The Breadth of Symplectic and Poisson Geometry: Festschrift in Honor of Alan Weinstein

The Breadth of Symplectic and Poisson Geometry Festschrift in Honor of Alan Weinstein Jerrold E. Marsden Tudor S. Ratiu...

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The Breadth of Symplectic and Poisson Geometry Festschrift in Honor of Alan Weinstein

Jerrold E. Marsden Tudor S. Ratiu Editors

Birkhäuser Boston • Basel • Berlin

Jerrold E. Marsden California Institute of Technology Department of Engineering and Applied Science Control and Dynamical Systems Pasadena, CA 91125 U.S.A.

Tudor S. Ratiu Ecole Polytechnique Fédérale de Lausanne Département de Mathématiques CH-1015 Lausanne Switzerland

AMS Subject Classifications: 53Dxx, 17Bxx, 22Exx, 53Dxx, 81Sxx Library of Congress Cataloging-in-Publication Data The breadth of symplectic and Poisson geometry : festschrift in honor of Alan Weinstein / Jerrold E. Marsden, Tudor S. Ratiu, editors. p. cm. – (Progress in mathematics ; v. 232) Includes bibliographical references and index. ISBN 0-8176-3565-3 (acid-free paper) 1. Symplectic geometry. 2. Geometric quantization. 3. Poisson manifolds. I. Weinstein, Alan, 1943- II. Marsden, Jerrold E. III. Ratiu, Tudor S. IV. Progress in mathematics (Boston, Mass.); v. 232. QA665.B74 2004 516.3’.6-dc22

ISBN 0-8176-3565-3

2004046202

Printed on acid-free paper.

c 2005 Birkhäuser Boston

All rights reserved. This work may not be translated or copied in whole or in part without the written permission of the publisher (Birkhäuser Boston, c/o Springer Science+Business Media Inc., Rights and Permissions, 233 Spring Street, New York, NY 10013, USA), except for brief excerpts in connection with reviews or scholarly analysis. Use in connection with any form of information storage and retrieval, electronic adaptation, computer software, or by similar or dissimilar methodology now known or hereafter developed is forbidden. The use in this publication of trade names, trademarks, service marks and similar terms, even if they are not identified as such, is not to be taken as an expression of opinion as to whether or not they are subject to proprietary rights. Printed in the United States of America. 987654321 www.birkhauser.com

SPIN 10958261

(JLS/HP)

Margo, Alan, and Asha in Paris at the lovely Fontaine des Quatre Parties du Monde.

Contents

Preface . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . ix Academic genealogy of Alan Weinstein . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xiii About Alan Weinstein . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xv Students of Alan Weinstein . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xv Alan Weinstein’s publications . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xvi Dirac structures, momentum maps, and quasi-Poisson manifolds Henrique Bursztyn, Marius Crainic . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . .

1

Construction of Ricci-type connections by reduction and induction Michel Cahen, Simone Gutt, Lorenz Schwachhöfer . . . . . . . . . . . . . . . . . . . . . . . 41 A mathematical model for geomagnetic reversals J. J. Duistermaat . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 59 Nonholonomic systems via moving frames: Cartan equivalence and Chaplygin Hamiltonization Kurt Ehlers, Jair Koiller, Richard Montgomery, Pedro M. Rios . . . . . . . . . . . . . 75 Thompson’s conjecture for real semisimple Lie groups Sam Evens, Jiang-Hua Lu . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 121 The Weinstein conjecture and theorems of nearby and almost existence Viktor L. Ginzburg . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 139 Simple singularities and integrable hierarchies Alexander B. Givental, Todor E. Milanov . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 173 Momentum maps and measure-valued solutions (peakons, filaments, and sheets) for the EPDiff equation Darryl D. Holm, Jerrold E. Marsden . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 203

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Higher homotopies and Maurer–Cartan algebras: Quasi-Lie–Rinehart, Gerstenhaber, and Batalin–Vilkovisky algebras Johannes Huebschmann . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 237 Localization theorems by symplectic cuts Lisa Jeffrey, Mikhail Kogan . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 303 Refinements of the Morse stratification of the normsquare of the moment map Frances Kirwan . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 327 Quasi, twisted, and all that… in Poisson geometry and Lie algebroid theory Yvette Kosmann-Schwarzbach . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 363 Minimal coadjoint orbits and symplectic induction Bertram Kostant . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 391 Quantization of pre-quasi-symplectic groupoids and their Hamiltonian spaces Camille Laurent-Gengoux, Ping Xu . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 423 Duality and triple structures Kirill C. H. Mackenzie . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 455 Star exponential functions as two-valued elements Y. Maeda, N. Miyazaki, H. Omori, A. Yoshioka . . . . . . . . . . . . . . . . . . . . . . . . . . 483 From momentum maps and dual pairs to symplectic and Poisson groupoids Charles-Michel Marle . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 493 Construction of spectral invariants of Hamiltonian paths on closed symplectic manifolds Yong-Geun Oh . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 525 The universal covering and covered spaces of a symplectic Lie algebra action Juan-Pablo Ortega, Tudor S. Ratiu . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 571 Poisson homotopy algebra: An idiosyncratic survey of homotopy algebraic topics related to Alan’s interests Jim Stasheff . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 583 Dirac submanifolds of Jacobi manifolds Izu Vaisman . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 603 Quantum maps and automorphisms Steve Zelditch . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 623

Preface

Alan Weinstein is one of the top mathematicians in the world working in the area of symplectic and differential geometry. His research on symplectic reduction, Lagrangian submanifolds, groupoids, applications to mechanics, and related areas has had a profound influence on the field. This area of research remains active and vibrant today and this volume is intended to be a reflection of that vigor. In addition to reflecting the vitality of the field, this is a celebratory volume to honor Alan’s 60th birthday. His birthday was also celebrated in August, 2003 with a wonderful week-long conference held at the ESI: the Erwin Schrödinger International Institute for Mathematical Physics in Vienna. Alan was born in New York in 1943. He was an undergraduate at MIT and a graduate student at UC Berkeley, where he was awarded his Ph.D. in 1967 under the direction of S. S. Chern. After spending postdoctoral years at IHES near Paris, MIT, and the University of Bonn, he joined the faculty at UC Berkeley in 1969, becoming a full Professor in 1976. Alan has received many honors, including an Alfred P. Sloan Foundation Fellowship, a Miller Professorship (twice), a Guggenheim Fellowship, election to the American Academy of Arts and Sciences in 1992, and an honorary degree at the University of Utrecht in 2003. At the ESI conference, S. S. Chern, Alan’s advisor, sent the following words to celebrate the occasion: “I am glad about this celebration and I think Alan richly deserves it. Alan came to me in the early sixties as a graduate student at the University of California at Berkeley. At that time, a prevailing problem in our geometry group, and the geometry community at large, was whether on a Riemannian manifold the cut locus and the conjugate locus of a point can be disjoint. Alan immediately showed that this was possible. The result became part of his Ph.D. thesis, which was published in the Annals of Mathematics. He received his Ph.D. degree in a short period of two years. I introduced him to IHES and the French mathematical community. He stays close with them and with the mathematical ideas of Charles Ehresmann. He is original and

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often came up with ingenious ideas. An example is his contribution to the solution of the Blaschke conjecture. I am very proud to count him as one of my students and I hope he will remain interested in mathematics up to my age, which is now 91.’’ Alan’s technical contributions are wide ranging and deep. As many of his early papers in his publication list illustrate, he started off in his thesis and the years immediately following in pure differential geometry, a topic he has come back to from time to time throughout his career. Already starting with his postdoc years and his early career at Berkeley, he became interested in symplectic geometry and mechanics. In this area he rapidly established himself as one of the world’s authorities, producing important and deep results ranging from reduction theory to Lagrangian and Poisson manifolds to studies of periodic orbits in Hamiltonian systems. He also did important work in fluid mechanics and plasma physics and through this work, he established warm relations with the Berkeley physicists Allan Kaufman and Robert Littlejohn. Alan’s important work on periodic orbits in Hamiltonian systems led him eventually to formulate the “Weinstein conjecture,’’ namely that for a given Hamiltonian flow on a symplectic manifold, there must be at least one closed orbit on a regular compact contact type level set of the Hamiltonian. Along with Arnold’s conjecture, the Weinstein conjecture has been one of the driving forces in symplectic topology over the last two decades. Alan kept up his interest in symplectic reduction theory throughout his later work. For instance, he laid some important foundation stones in the theory of semidirect product reduction as well as in singular reduction through his work on Satake’s V -manifolds, along with finding important links with singular structures in moduli spaces. Intertwined with his work on symplectic geometry and mechanics, he did extensive work on geometric PDE, eigenvalues, the Schrödinger operator and geometric quantization. Alan took the point of view of microlocal analysis and phase space structures in his work in this area, emphasizing the links with quantum mechanics.

Preface

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His work on the limit distribution of eigenvalue clusters in terms of the geodesic Radon transform of the potential inspired a large number of related articles. He showed that the geodesic flow of a Zoll surface was symplectically equivalent to that of a round sphere, and hence that its Laplacian could be conjugated globally to the round Laplacian plus a pseudodifferential potential. This work inspired many other results on conjugacies. One of Alan’s fundamental contributions to Poisson geometry was the introduction of symplectic groupoids in 1987, which marks the official beginning of his “oids’’ period. In these works, he makes sweeping generalizations about a wide variety of constructions in symplectic geometry, including (with Courant) the important notion of Dirac structures. During this period of generalizations he constantly returned to specific topics in symplectic and Poisson geometry, such as geometric phases and Poisson Lie groups, in addition to making other key links. For instance, symplectic groupoids are used to link Poisson geometry to noncommutative geometry, and groupoids are also intimately related to many other areas, including symmetries and reduction, dual pairs, quantization and the theory of sigma models. One of the central ideas is that the usual theory of Hamiltonian actions, momentum maps, and symplectic reduction makes sense in the more general context of actions of symplectic groupoids; in this setting, momentum maps are Poisson maps taking values in general Poisson manifolds, rather than just Lie–Poisson manifolds (that is, duals of Lie algebras). Alan has raised the question of whether this framework can be further extended to include new notions of momentum maps such as quasi-Poisson manifolds with group-valued momentum maps as well as optimal momentum maps. Alan is well known not only for his brilliant papers and conjectures, but also for his general philosophy, such as the symplectic creed: Everything is a Lagrangian submanifold . Those of us who know him well also appreciate his very special insight. For example, in the middle of a discussion (for instance, as we both had in our joint works on semidirect product reduction as well as stability theory) he will say something like what you are really doing is. . . and then give us some usually very special insight that invariably substantially improves the whole project. Alan also has a very interesting and charming sense of humor that even makes its way into his papers from time to time. For instance, Alan had great fun in his papers with the “East Coast–West Coast’’ discussions of whether one should use the term momentum map or moment map. He also gave us a good laugh with the term symplectic bones as it relates to the French translation of Poisson as Fish. Alan is a great educator. His lectures, even on Calculus, are always a treat and are very inspiring for their special insight, their wit and lively presentation. His enthusiasm for mathematics is infectious. One story that comes to mind on the education front is this: during the days when he was exceptionally keen about groupoids, he was preparing a lecture for undergraduates on the subject. Some of us convinced him to present it as a colloquium lecture for faculty, keeping in mind the old advice “no colloquium talk can be too simple.’’ It was, in fact, not only a beautiful colloquium talk, but was perfectly pitched for the faculty, and it became a popular article in the Notices of the American Mathematical Society. Part of being a good educator is being

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cognizant of history. Alan excels in this area. For instance, his research into the history of Lie is what led directly to the introduction of the term “Lie–Poisson’’ bracket. The papers in this volume were selected by invitation and all of them underwent a rigorous refereeing process. While this process took some time, it resulted in high quality papers. We thank all of the referees for their diligent and helpful work. The authors of this volume represent some of the best workers in the subject and their contributions span a wide range of the topics covered by symplectic and Poisson geometry and mechanics, broadly interpreted. The intended audience for the book includes active researchers in the general area of symplectic geometry and mechanics, as well as aspiring graduate students who wish to learn where the subject is headed and what some of the current research topics are. Alan and Margo have a special relationship to Paris. They have spent many happy times there, and we wish them all the best and many more happy visits in the years to come. We wish to thank Ann Kostant for her expert editorial guidance throughout the production of this volume. Of course, we also thank all the authors for their contributions as well as their helpful guidance and advice. The referees are also thanked for their valuable comments and suggestions.

Jerry Marsden and Tudor Ratiu September, 2004

Academic genealogy of Alan Weinstein

Otto Mencken Universität Leipzig, 1668 Thomae Hobbesii Epicureismum historice delineatum sistit Johann C. Wichmannshausen Universität Leipzig, 1685 Disputationem Moralem De Divortiis Secundum Jus Naturae Christian A. Hausen Martin-Luther-Universität Halle-Wittenberg, 1713 De corpore scissuris figurisque non cruetando ductu Abraham G. Kaestner Universität Leipzig, 1739 Theoria radicum in aequationibus Johann F. Pfaff Georg-August-Universität Gottingen, 1786 Commentatio de ortibus et occasibus siderum apud auctores classicos commemoratis August F. Möbius Universität Leipzig, 1815 De computandis occultationibus fixarum per planetas Otto W. Fiedler Universität Leipzig, 1859

Johannes Frischauf Universität Wien, 1861

Karl Friesach Universität Wien, 1846

Gustav Ritter von Escherich Technische Universität Graz, 1873 Die Geometrie auf Flachen constanter negativer Krummung

Emil Weyr University of Prague, 1870

Wilhelm Wirtinger Universität Wien, 1887 Uber eine spezielle Tripelinvolution in der Ebene

Wilhelm Blaschke Universität Wien, 1908 Shiing-Shen Chern Universität Hamburg, 1936 Eine Invariantentheorie der Dreigewebe aus r-dimensionalen Mannigfaltigkeiten im R2r Alan D. Weinstein University of California at Berkeley, 1967 The Cut Locus and Conjugate Locus of a Riemannian Manifold

About Alan Weinstein

Alan David Weinstein Ph.D.: University of California at Berkeley, 1967 Dissertation: The Cut Locus and Conjugate Locus of a Riemannian Manifold Advisor: Shiing-Shen Chern

Students of Alan Weinstein 1. 2. 3. 4. 5. 6. 7. 8. 9. 10. 11. 12. 13. 14. 15.

Jair Koiller, Studies on the Spring-Pendulum, 1975 Otto Ruiz, Existence of Brake-Orbits in Finsler Mechanical Systems, 1975 Yilmaz Akyildiz, Dynamical Symmetries of the Kepler Problem, 1976 Gerald Chachere, Numerical Experiments Concerning the Eigenvalues of the Laplacian on a Zoll Surface, 1977 John Jacob, Geodesic Symmetries of Homogeneous Kahler Manifolds, 1977 Steven Zelditch, Reconstruction of Singularities for Solutions of Schrödinger’s Equations, 1981 Enrique Planchart, Analogies in Symplectic Geometry of Some Results of Cartan in Representation Theory, 1982 Barry Fortune, A Symplectic Fixed Point Theorem for Complex Projective Spaces, 1984 Stephen Omohundro (Department of Physics), Geometric Perturbation Theory in Physics, 1985 Theodore Courant, Dirac Manifolds, 1987 Yong-Geun Oh, Nonlinear Schrödinger Equations with Potentials: Evolution, Existence, and Stability of Semi-Classical Bound States, 1988 Viktor Ginzburg, On Closed Characteristics of 2-Forms, 1990 Milton Lopes Filho, Microlocal Regularity and Symbols for Distributions, 1990 Jiang-Hua Lu, Multiplicative and Affine Poisson Structures on Lie Groups, 1990 Ping Xu, Morita Equivalence of Poisson Manifolds, 1990

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16. Sean Bates, Symplectic End Invariants and C 0 Symplectic Topology, 1994 17. Agust Egilsson, On Embedding a Stratified Symplectic Space in a Smooth Poisson Manifold , 1995 18. Dong Yan, Yang–Mills Theory on Symplectic Manifolds, 1995 19. Zhao-Hui Qian, Groupoids, Midpoints and Quantizations, 1997 20. Vinay Kathotia, Universal Formulae for Deformation Quantization and The Campbell–Baker–Hausdorff Formula, 1998 21. Dmitry Roytenberg, Courant Algebroids, Derived Brackets And Even Symplectic Supermanifolds, 1999 22. Mélanie Bertelson-Volckaert (Stanford University), Foliations Associated to Regular Poisson Structures, 2000 23. Benjamin Davis, On Poisson Spaces Associated to Finitely Generated Poisson R-Algebras, 2001 24. Henrique Bursztyn, Morita Equivalence in Deformation Quantization, 2001 25. Olga Radko, Some Invariants of Poisson Manifolds, 2002 26. Xiang Tang, Quantization of Noncommutative Poisson Manifolds, 2003 27. Marco Zambon, Submanifold Averaging in Riemannian, Symplectic, and Contact Geometry, 2003 28. Chenchang Zhu, Integrating Lie Algebroids via Stacks and Applications to Jacobi Manifolds, 2003

Alan Weinstein’s publications [1] Weinstein, A., On the homotopy type of positively pinched manifolds, Arch. Math., 18 (1967), 523–524. [2] Weinstein, A., A fixed point theorem for positively curved manifolds, J. Math. Mech., 18 (1968), 149–153. [3] Weinstein, A., The cut locus and conjugate locus of a riemannian manifold, Ann. Math. 87 (1968), 29–41. [4] Weinstein, A., Symplectic structures on Banach manifolds, Bull. Amer. Math. Soc., 75 (1969), 1040–1041. [5] Weinstein, A., and Simon, U., Anwendungen der de rhamschen Zerlegung auf Probleme der localen Flächentheorie, Manuscripta Math., 1 (1969), 139–146. [6] Marsden, J., and Weinstein, A., A comparison theorem for hamiltonian vector fields, Proc. Amer. Math. Soc., 26 (1970), 629–631. [7] Weinstein,A., The generic conjugate locus, in Global Analysis, Proceedings of Symposia on Pure Mathematics, Vol. 15, American Mathematical Society, Providence, RI, 1970, 299–301. [8] Weinstein, A., Positively curved n-manifolds in R n+2 , J. Differential Geom., 4 (1970), 1–4. [9] Weinstein, A., Positively curved deformations of invariant Riemannian metrics, Proc. Amer. Math. Soc., 26 (1970), 151–152. [10] Weinstein, A., Sur la non-densité des géodésiques fermées, C. R. Acad. Sci. Paris, 271 (1970), 504. [11] Roels, J., and Weinstein, A., Functions whose Poisson brackets are constants, J. Math. Phys., 12 (1971), 1482–1486.


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[12] Weinstein, A., Singularities of families of functions, in Proceedings of the Conference “Differentialgeometrie im Grossen,’’ Mathematische Forschungsinstitut, Oberwolfach, Germany, 1971, 323–330. [13] Weinstein, A., Perturbation of periodic manifolds of Hamiltonian systems, Bull. Amer. Math. Soc., 77 (1971), 814–818. [14] Weinstein, A., Remarks on curvature and the Euler integrand, J. Differential Geom., 6 (1971), 259–262. [15] Weinstein, A., Symplectic manifolds and their lagrangian submanifolds, Adv. Math., 6 (1971), 329–346. [16] Weinstein, A., On the invariance of Poincaré’s generating function for canonical transformations, Invent. Math., 16 (1972), 202–213. [17] Weinstein, A., Distance spheres in complex projective spaces, Proc. Amer. Math. Soc., 39 (1973), 649–650. [18] Weinstein, A., Lagrangian submanifolds and hamiltonian systems, Ann. Math., 98 (1973), 377–410. [19] Weinstein, A., Normal modes for nonlinear hamiltonian systems, Invent. Math., 20 (1973), 47–57. [20] Marsden, J., and Weinstein, A., Reduction of symplectic manifolds with symmetry, Rep. Math. Phys., 5 (1974), 121–130. [21] Weinstein, A., Application des opérateurs intégraux de Fourier aux spectres des variétés riemanniennes, C. R. Acad. Sci. Paris, 279 (1974), 229–230. [22] Weinstein, A., On the volume of manifolds, all of whose geodesics are closed, J. Differential Geom., 9 (1974), 513–517. [23] Weinstein, A., Quasi-classical mechanics on spheres, Sympos. Math., 14 (1974), 25–32. [24] Weinstein, A., On Maslov’s quantization condition, in Proceedings of the International Symposium on Fourier Integral Operators (Nice, May 1974), Lecture Notes in Mathematics, Vol. 469, Springer-Verlag, New York, 1975, 341–372. [25] Guillemin, V., and Weinstein, A., Eigenvalues associated with a closed geodesic, Bull. Amer. Math. Soc., 82 (1976), 92–94. [26] Weinstein, A., Fourier integral operators, quantization, and the spectrum of a Riemannian manifold, in Géométrie Symplectique et Physique Mathématique, Colloque Internationale de Centre National de la Recherche Scientifique No. 237, CNRS, Paris, 1976, 289–298. [27] Weinstein, A., The principal symbol of a distribution, Bull. Amer. Math. Soc., 82 (1976), 548–550. [28] Weinstein, A., Symplectic V -manifolds, periodic orbits of Hamiltonian systems, and the volume of certain Riemannian manifolds, Comm. Pure Appl. Math., 30 (1977), 265–271. [29] Weinstein, A., Lectures on Symplectic Manifolds, Regional Conference Series in Mathematics, Vol. 29, American Mathematical Society, Providence, RI, 1977. [30] Weinstein, A., Asymptotics of eigenvalue clusters for the Laplacian plus a potential, Duke Math. J., 44 (1977), 883–892. [31] Weinstein, A., The order and symbol of a distribution, Trans. Amer. Math. Soc., 241 (1978), 1–54. [32] Weinstein, A., Simple periodic orbits, Amer. Inst. Phys. Conf. Proc., 46 (1978), 260–263. [33] Weinstein, A., Eigenvalues of the laplacian plus a potential, in Proceedings of the International Congress of Mathematicians, Helsinki, 1978, 803–805. [34] Weinstein, A., A universal phase space for particles in Yang–Mills fields, Lett. Math. Phys., 2 (1978), 417–420. [35] Weinstein, A., Periodic orbits for convex hamiltonian systems, Ann. Math., 108 (1978), 507–518.

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[36] Weinstein, A., Bifurcations and Hamilton’s principle, Math. Z., 159 (1978), 235–248. [37] Weinstein, A., On the hypotheses of Rabinowitz’ periodic orbit theorems, J. Differential Equations 33 (1979), 353–358. [38] Marsden, J. E., and Weinstein, A., Review of Geometric Asymptotics and Symplectic Geometry and Fourier Analysis, Bull. Amer. Math. Soc., 1 (1979), 545–553. [39] Marsden, J., and Weinstein, A., Calculus, Benjamin/Cummings, San Francisco, 1980. [40] Weinstein, A., Fat bundles and symplectic manifolds, Adv. Math., 37 (1980), 239–250. [41] Weinstein, A., Nonlinear stabilization of quasimodes, in Proceedings of the AMS Symposium on Geometry of the Laplacian, Hawaii, 1979, Proceedings of Symposia on Pure Mathematics, Vol. 36, American Mathematical Society, Providence, RI, 1980, 301–318. [42] Marsden, J., and Weinstein, A., Calculus Unlimited , Benjamin/Cummings, San Francisco, 1981. [43] Croke, C., and Weinstein, A., Closed curves on convex hypersurfaces and periods of nonlinear oscillations, Invent. Math., 64 (1981), 199–202. [44] Marsden, J., Morrison, P., and Weinstein, A., Comments on: The Maxwell–Vlasov equations as a continuous Hamiltonian system, Phys. Lett., 96A (1981), 235–236. [45] Stanton, R. J., and Weinstein A., On the L4 norm of spherical harmonics, Math. Proc. Cambridge Philos. Soc., 89 (1981), 343–358. [46] Weinstein, A., Symplectic geometry, Bull. Amer. Math. Soc. (N.S.), 5 (1981), 1–13. [47] Weinstein, A., Neighborhood classification of isotropic embeddings, J. Differential Geom., 16 (1981), 125–128. [48] Marsden. J., and Weinstein, A., The hamiltonian structure of the Maxwell–Vlasov equations, Physica, 4D (1982), 394–406. [49] Weinstein, A., Gauge groups and Poisson brackets for interacting particles and fields, Amer. Inst. Phys. Conf. Proc., 88 (1982), 1–11. [50] Weinstein, A., What is microlocal analysis?, Math. Intel., 4 (1982), 90–92. [51] Weinstein, A., The symplectic “category,’’ in Doebner, H.-D., Andersson, S. I., and Petry, H. R., eds., Differential Geometric Methods in Mathematical Physics (Clausthal, Germany 1980), Lecture Notes in Mathematics, Vol. 905, Springer-Verlag, Berlin, 1982, 45–50. [52] Weinstein, A., and Zelditch, S., Singularities of solutions of some Schrödinger equations on R n , Bull. Amer. Math. Soc., (1982). [53] Gotay, M. J., Lashof, R., Sniatycki, J., and Weinstein, A., Closed forms on symplectic fibre bundles, Comm. Math. Helv., 58 (1983), 617–621. [54] Marsden, J., Ratiu, T., Schmid, R., Spencer, R., and Weinstein, A., Hamiltonian systems with symmetry, coadjoint orbits, and plasma physics, Atti Acad. Sci. Torino, 117Supplemento (1983), 289–340. [55] Marsden, J., and Weinstein, A., Coadjoint orbits, vortices and Clebsch variables for incompressible fluids, Physica, 7D (1983), 305–323. [56] Sniatycki, J., and Weinstein, A., Reduction and quantization for singular momentum mappings, Lett. Math. Phys., 7 (1983), 159–161. [57] Weinstein, A., A symplectic rigidity theorem, Duke Math. J., 50 (1983), 1121–1125. [58] Weinstein, A., Hamiltonian structure for drift waves and geostrophic flow, Phys. Fluids, 26, (1983), 388–390. [59] Weinstein, A., Sophus Lie and symplectic geometry, Expos. Math., 1 (1983), 95–96. [60] Weinstein, A., Removing intersections of lagrangian immersions, Illinois J. Math., 27 (1983), 484–500. [61] Weinstein, A., The local structure of Poisson manifolds, J. Differential Geom., 18 (1983), 523–557.


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[62] Marsden, J., Morrison, P., and Weinstein, A., The Hamiltonian structure of the BBGKY hierarchy equations, Contemp. Math., 28 (1984), 115–124. [63] Marsden, J., Ratiu, T., and Weinstein, A., Reduction and Hamiltonian structures on duals of semidirect product Lie algebras, Contemp. Math., 28 (1984), 55–100. [64] Marsden. J., Ratiu, T., and Weinstein, A., Semidirect products and reduction in mechanics, Trans. Amer. Math. Soc., 281 (1984), 147–177. [65] Weinstein, A., Equations of plasma physics (notes by Stephen Omohundro), in Chern, S. S., ed., Seminar on Nonlinear Partial Differential Equations, MSRI Publications, Springer-Verlag, New York, 1984, 359–373. [66] Weinstein, A., Stability of Poisson-Hamiltonian equilibria, Contemp. Math., 28 (1984), 3–13. [67] Weinstein, A., C 0 perturbation theorems for symplectic fixed points and lagrangian intersections, Travaux en Cours, 3 (1984), 140–144. [68] Fortune, B., and Weinstein, A., A symplectic fixed point theorem for complex projective spaces, Bull. Amer. Math. Soc., 12 (1985), 128–130. [69] Holm. D. D., Marsden, J. E., Ratiu, T., and Weinstein, A., Nonlinear stability of fluid and plasma equilibria, Phys. Rep., 123-1–2 (1985), 1–116. [70] Marsden, J., and Weinstein, A., Calculus I, II, III, 2nd ed., Springer-Verlag, New York, 1985. [71] Weinstein, A., A symbol calculus for some Schrödinger equations on R n , Amer. J. Math., (1985), 1–21. [72] Weinstein, A., A global invertibility theorem for manifolds with boundary, Proc. Roy. Soc. Edinburgh Sect. A, 99 (1985), 283–284. [73] Weinstein, A., Periodic nonlinear waves on a half-line, Comm. Math. Phys., 99 (1985), 385–388. [74] Weinstein, A., Poisson structures and Lie algebras, Astérisque, hors série (1985), 421– 434. [75] Weinstein, A., Symplectic reduction and fixed points, in Séminaire Sud-Rhodanien de Géométrie, Rencontre de Balaruc I, Travaux en Cours, Hermann, Paris, 1985, 140–148. [76] Weinstein, A., Three dimensional contact manifolds with vanishing torsion tensor (appendix to a paper by S. S. Chern and R. Hamilton), in Hirzebruch, F., Schwermer J., and Suter S., eds., Proceedings of the Meeting held by the Max-Planck-Institut für Mathematik, Bonn. June 15–22, 1984, Lecture Notes in Mathematics, Vol. 1111, SpringerVerlag, Berlin, 1985, 306–308. [77] Floer, A., and Weinstein A., Nonspreading wave packets for the nonlinear Schrödinger equation with a bounded potential, J. Functional Anal., 69 (1986), 397–408. [78] Weinstein, A., On extending the Conley-Zehnder theorem to other manifolds, Proc. Sympos. Pure Math., 45 (1986), 541–544. [79] Weinstein, A., Critical point theory, symplectic geometry, and hamiltonian systems, in Proceedings of the 1983 Beijing Symposium on Differential Geometry and Differential Equations, Science Press, Beijing, 1986, 261–289. [80] Coste, A., Dazord, P., and Weinstein, A., Groupoïdes symplectiques, Publ. Dép. Math. Univ. Claude Bernard-Lyon I, 2A (1987), 1–62. [81] Weinstein, A., ed., Some Problems in Symplectic Geometry, Séminaire Sud-Rhodanien de Géométrie VI, Travaux en Cours, Hermann, Paris, 1987. [82] Weinstein, A., Standing and travelling waves for nonlinear wave equations, Transport Theory Stat. Phys., 16 (1987), 267–277. [83] Weinstein, A., The Geometry of Poisson Brackets (Notes by K. Ono and K. Sugiyama), Surveys in Geometry, Tokyo, 1987.

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[84] Weinstein, A., Poisson geometry of the principal series and nonlinearizable structures, J. Differential Geom., 25 (1987), 55–73. [85] Weinstein, A., Symplectic groupoids and Poisson manifolds, Bull. Amer. Math. Soc., 16, (1987), 101–104. [86] Courant, T. J., and Weinstein, A., Beyond Poisson structures, in Séminaire SudRhodanien de Géométrie VIII, Travaux en Cours, Vol. 27, Hermann, Paris, 1988, 39–49. [87] Mikami, K., and Weinstein, A., Moments and reduction for symplectic groupoid actions, Publ. RIMS Kyoto Univ., 24 (1988), 121–140. [88] Weinstein, A., Coisotropic calculus and Poisson groupoids, J. Math. Soc. Japan, 40 (1988), 705–727. [89] Weinstein, A., Some remarks on dressing transformations, J. Fac. Sci. Univ. Tokyo. Sect. 1A Math., 36 (1988), 163–167. [90] Lu, J.-H., and Weinstein, A., Groupoïdes symplectiques doubles des groupes de LiePoisson, C. R. Acad. Sci. Paris, 309 (1989), 951–954. [91] Weinstein, A., Cohomology of symplectomorphism groups and critical values of hamiltonians, Math. Z., 201 (1989), 75–82. [92] Weinstein, A., Blowing up realizations of Heisenberg–Poisson manifolds, Bull. Sci. Math., 113 (1989), 381–406. [93] Lu, J.-H., and Weinstein, A., Poisson Lie groups, dressing transformations, and the Bruhat decomposition, J. Differential Geom., 31 (1990), 501–526. [94] Weinstein, A., Connections of Berry and Hannay type for moving lagrangian submanifolds, Adv. Math., 82 (1990), 133–159. [95] Weinstein, A., Affine Poisson structures, Internat. J. Math., 1 (1990), 343–360. [96] Dazord, P., Lu, J.-H., Sondaz, D., and Weinstein, A., Affinoïdes de Poisson, C. R. Acad. Sci. Paris, 312 (1991), 523–527. [97] Hofer, H., Weinstein, A., and Zehnder, E., Andreas Floer, 1956–1991 (obituary), Notices Amer. Math. Soc., 38 (1991), 910–911. [98] Lu, J.-H., and Weinstein, A., Classification of SU (2)-covariant Poisson structures on S 2 (appendix to a paper of A. J.-L. Sheu), Comm. Math. Phys., 135 (1991), 229–232. [99] Weinstein, A., Symplectic groupoids, geometric quantization, and irrational rotation algebras, in Symplectic Geometry, Groupoids, and Integrable Systems: Séminaire SudRhodanien de Géométrie à Berkeley (1989), Dazord, P., and Weinstein, A., eds., Springer–MSRI Series, Springer-Verlag, New York, 1991, 281–290. [100] Weinstein, A., Contact surgery and symplectic handlebodies, Hokkaido Math. J., 20 (1991), 241–251. [101] Weinstein, A., Noncommutative geometry and geometric quantization, in Donato, P., Duval, C., Elhadad, J., and Tuynman, G. M., eds., Symplectic Geometry and Mathematical Physics: Actes du Colloque en l’Honneur de Jean-Marie Souriau, Progress in Mathematics, Birkhäuser, Basel, 1991, 446–461. [102] Weinstein, A., and Xu, P., Extensions of symplectic groupoids and quantization, J. Reine Angew. Math., 417 (1991), 159–189. [103] Ginzburg, V. L., and Weinstein, A., Lie–Poisson structure on some Poisson Lie groups, J. Amer. Math. Soc., 5 (1992), 445–453. [104] Weinstein, A., and Xu, P., Classical solutions of the quantum Yang–Baxter equation, Comm. Math. Phys., 148 (1992), 309–343. [105] Mardsen, J. E., Tromba,A. J., and Weinstein,A., Basic Multivariable Calculus, SpringerVerlag and W. H. Freeman, New York, 1993. [106] Weinstein, A., Traces and triangles in symmetric symplectic spaces, Contemp. Math., 179 (1994), 261–270.


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[107] Maeda, Y., Omori, H., and Weinstein, A., eds., Symplectic Geometry and Quantization: Two Symposia on Symplectic Geometry and Quantization Problems, July 1993, Japan, Contemporary Mathematics, Vol. 179, American Mathematical Society, Providence, RI, 1994. [108] Weinstein, A., Classical theta functions and quantum tori, Publ. RIMS Kyoto Univ., 30 (1994), 327–333. [109] Birnir, B., McKean, H., and Weinstein, A., The rigidity of sine-Gordon breathers, Comm. Pure Appl. Math., 47 (1994), 1043–1051. [110] Scovel, C., and WeinsteinA., Finite dimensional Lie–Poisson approximations to Vlasov– Poisson equations, Comm. Pure Appl. Math., 47 (1994), 683–709. [111] Emmrich, C., and Weinstein, A., The differential geometry of Fedosov’s quantization, in Brylinski, J. L., Brylinski, R., Guillemin, V., and Kac, V., eds., Lie Theory and Geometry: In Honor of B. Kostant, Progress in Mathematics, Birkhäuser, Boston, 1994, 217–239. [112] Weinstein, A., Deformation quantization, Astérisque, 227 (1995) (Séminaire Bourbaki, 46ème année, 1993–94, no. 789), 389–409. [113] Bates, S., and Weinstein, A., Lectures on the Geometry of Quantization, Berkeley Mathematics Lecture Notes, American Mathematical Society, Providence, RI, 1997. [114] Weinstein, A., The symplectic structure on moduli space, in Hofer, H., Taubes, C., Weinstein, A., and Zehnder, E., eds., The Floer Memorial Volume, Birkhäuser, Basel, 1995, 627–635. [115] Weinstein, A., Lagrangian mechanics and groupoids, in Shadwick, W. F., Krishnaprasad, P. S., and Ratiu, T. S., eds., Mechanics Day, Fields Institute Communications, Vol. 7., American Mathematical Society, Providence, RI, 1995, 207–231. [116] Emmrich, C., and Weinstein, A., Geometry of the transport equation in multicomponent WKB approximations, Comm. Math. Phys., 176 (1996), 701–711. [117] Weinstein, A., Groupoids: Unifying internal and external symmetry, Notices Amer. Math. Soc., 43 (1996), 744–752; reprinted in Contemp. Math., 282 (2001), 1–19. [118] Reshetikhin, N., Voronov, A. A., and Weinstein, A., Semiquantum geometry, Algebraic geometry 5, J. Math. Sci., 82 (1996), 3255–3267. [119] Guruprasad, K., Huebschmann, J., Jeffrey, L., and Weinstein, A., Group systems, groupoids, and moduli spaces of parabolic bundles, Duke Math. J., 89 (1997), 377– 412. [120] Weinstein, A., Tangential deformation quantization and polarized symplectic groupoids, in Gutt, S., Rawnsley, J., and Sternheimer, D., eds., Deformation Theory and Symplectic Geometry, Mathematical Physics Studies, Vol. 20, Kluwer, Dordrecht, the Netherlands, 1997, 301–314. [121] Liu, Z.-J., Weinstein, A., and Xu, P., Manin triples for Lie bialgebroids, J. Differential Geom., 45 (1997), 547–574. [122] Weinstein, A., The modular automorphism group of a Poisson manifold, J. Geom. Phys., 23 (1997), 379–394. [123] Weinstein, A., Some questions about the index of quantized contact transformations, RIMS Kôkyûroku, 1014 (1997), 1–14. [124] Weinstein, A., and Xu, P., Hochschild cohomology and characteristic classes for starproducts, in Khovanskii, A., Varchenko, A., and Vassiliev, V., eds., Geometry of Differential Equations, American Mathematical Society, Providence, RI, 1997, 177–194. [125] Liu, Z.-J., Weinstein, A., and Xu, P., Dirac structures and Poisson homogeneous spaces, Comm. Math. Phys., 192 (1998), 121–144. [126] Weinstein, A., Poisson geometry, Differential Geom. Appl., 9 (1998), 213–238. [127] Roytenberg, D., and Weinstein, A., Courant algebroids and strongly homotopy Lie algebras, Lett. Math. Phys., 46 (1998), 81–93.

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[128] Weinstein, A., From Riemann Geometry to Poisson Geometry and Back Again, Lecture at Chern Symposium, Mathematical Sciences Research Institute, Berkeley, CA, 1998; available from http://msri.org/publications/video/contents.html and on CD-ROM. [129] Cannas da Silva, A., and Weinstein, A., Geometric Models for Noncommutative Algebras, Berkeley Mathematics Lecture Notes, American Mathematical Society, Providence, RI, 1999. [130] Nistor, V., Weinstein, A., and Xu., P., Pseudodifferential operators on differential groupoids, Pacific J. Math. 189 (1999), 117–152. [131] Evens, S., Lu, J.-H., and Weinstein, A., Transverse measures, the modular class, and a cohomology pairing for Lie algebroids, Quart. J. Math., 50 (1999), 417–436. [132] Fuchs, D., Eliashberg, Y., Ratiu, T., and Weinstein, A., eds., Northern California Symplectic Geometry Seminar, American Mathematical Society, Providence, RI, 1999. [133] Weinstein, A., Almost invariant submanifolds for compact group actions, J. European Math. Soc., 2 (2000), 53–86. [134] Mikami, K., and Weinstein, A., Self-similarity of Poisson structures on tori, in Poisson Geometry, Banach Center Publications, Vol. 51, Polish Scientific Publishers PWN, Warsaw, 2000, 211–217. [135] Weinstein, A., Linearization problems for Lie algebroids and Lie groupoids, Lett. Math. Phys., 52 (2000), 93–102. [136] Weinstein, A., Omni-Lie algebras, RIMS Kôkyûroku, 1176 (2000), 95–102. [137] Weinstein, A., Review of Riemannian Geometry During the Second Half of the Twentieth Century by Marcel Berger, Bull. London Math. Soc., 33 (2001), 11. [138] Kinyon, M. K., and Weinstein, A., Leibniz algebras, Courant algebroids, and multiplications on reductive homogeneous spaces, Amer. J. Math., 123 (2001), 525–550. [139] Weinstein, A., Poisson geometry of discrete series orbits, and momentum convexity for noncompact group actions, Lett. Math. Phys., 56 (2001), 17–30. [140] Marsden, J., and Weinstein, A., Some comments on the history, theory, and applications of symplectic reduction, in Landsman, N. P., Pflaum, M., and Schlichenmaier, M., eds., Quantization of Singular Symplectic Quotients, Birkhäuser, Basel, 2001, 1–19. [141] Hirsch, M. W., and Weinstein, A., Fixed points of analytic actions of supersoluble Lie groups on compact surfaces, Ergodic Theory Dynam. Systems, 21 (2001), 1783–1787. [142] Ševera, P., and Weinstein, A., Poisson geometry with a 3-form background, Progr. Theoret. Phys. Suppl. Ser., 144 (2002), 145–154. [143] Weinstein, A., Linearization of regular proper groupoids, J. Inst. Math. Jussieu, 1 (2002), 493–511. [144] Newton, P. K., Holmes, P., and Weinstein,A., eds., Geometry, Mechanics, and Dynamics: Special Volume in Honor of the 60th Birthday of J. E. Marsden, Springer-Verlag, New York, 2002. [145] Bursztyn, H., and Weinstein, A., Picard groups in Poisson geometry, Moscow Math. J., 4 (2004), 39–66. [146] Weinstein, A., The geometry of momentum, in Proceedings of the Conference on “Geometry in the 20th Century: 1930–2000,’’ (Paris, September 2001), to appear; math.SG/0208108. [147] Bursztyn, H., Crainic, M., Weinstein, A., and Zhu, C., Integration of twisted Dirac brackets, Duke Math. J., 123 (2004), 549–607. [148] Tang, X., and Weinstein, A., Quantization and Morita equivalence for constant Dirac structures on tori, Ann. Inst. Fourier, 54 (2004), to appear; math.QA/0305413. [149] Weinstein, A., The Maslov gerbe, Lett. Math. Phys., to appear; math.SG/0312274.


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[150] Bursztyn, H., and Weinstein, A., Poisson geometry and Morita equivalence, in Poisson Geometry, Deformation Quantization, and Group Representations, London Mathematical Society Lecture Note Series, Cambridge University Press, Cambridge, UK, to appear; preprint math.SG/0402347. [151] Weinstein, A., Integrating the nonintegrable, in Proceedings of the Workshop “Feuilletages: Quantification Géométrique,’’ Maison des Science de l’Homme, Paris, 2004.

Dirac structures, momentum maps, and quasi-Poisson manifolds Henrique Bursztyn1 and Marius Crainic2 1 Department of Mathematics

University of Toronto Toronto, ON M5S 3G3 Canada [email protected] 2 Department of Mathematics Utrecht University P. O. Box 80.010, 3508 TA Utrecht The Netherlands [email protected] Dedicated to Alan Weinstein for his 60th birthday. Abstract. We extend the correspondence between Poisson maps and actions of symplectic groupoids, which generalizes the one between momentum maps and Hamiltonian actions, to the realm of Dirac geometry.As an example, we show how Hamiltonian quasi-Poisson manifolds fit into this framework by constructing an “inversion’’ procedure relating quasi-Poisson bivectors to twisted Dirac structures.

1 Introduction This paper builds on three ideas pursued by Alan Weinstein in some of his many fundamental contributions to Poisson geometry: First, Lie algebroids play a prominent role in the study of Poisson manifolds [8, 30]; second, Poisson maps can be regarded as generalized momentum maps for actions of symplectic groupoids [25, 31]; third, Poisson structures on manifolds are particular examples of more general objects called Dirac structures [12, 13, 28]. The main objective of this paper is to combine these three ideas in order to extend the notion of “momentum map’’ to the realm of Dirac geometry. As an application, we obtain an alternative approach to Hamiltonian quasi-Poisson manifolds [2] which answers many of the questions posed in [28, 31], shedding light on the relationship between various notions of generalized Poisson structures, Hamiltonian actions and reduced spaces. Let g be a Lie algebra, and consider its dual g∗ , equipped with its Lie–Poisson structure. The central ingredients in the formulation of classical Hamiltonian g-actions

2

H. Bursztyn and M. Crainic

are a Poisson manifold (Q, πQ ) and a Poisson map J : Q → g∗ , which we use to define an action of g on Q by Hamiltonian vector fields: g −→ X (Q),

v → XJv := idJv (πQ ),

(1.1)

where Jv ∈ C ∞ (Q) is given by Jv (x) = J (x), v. For the global picture, we assume that J is a complete Poisson map [8, Sec. 6.2], in which case the infinitesimal action (1.1) can be integrated to an action of the connected, simply connected Lie group G with Lie algebra g, in such a way that J becomes G-equivariant with respect to the coadjoint action of G on g∗ . The map J is called a momentum map for the G-action on Q, and we refer to the G-action as Hamiltonian. A key observation, described in [25, 31], is that this construction of a Hamiltonian action out of a Poisson map holds in much more generality: one may replace g∗ by any Poisson manifold, as long as Lie groups are replaced by symplectic groupoids [29]. In this sense, any Poisson map can be seen as a “Poisson-manifold valued moment map.’’ In this paper, we show that the correspondence between Poisson maps and Hamiltonian actions by symplectic groupoids can be further extended to the context of Dirac geometry: in this setting, Poisson maps must be replaced by special types of Dirac maps called Dirac realizations (see Definition 3.11); for the associated global actions, twisted presymplectic groupoids [6] (alternatively called quasi-symplectic groupoids [33]) play the role of symplectic groupoids. Our main results show that various important notions of generalized Hamiltonian actions, such as the “quasi’’ objects of [2, 3], fit nicely into the Dirac geometry framework. We organize our results as follows. In Section 2, we discuss important connections between Lie algebroids and bivector fields. Our main result is that, just as ordinary Poisson structures give rise to Lie algebroid structures on their cotangent bundles, a quasi-Poisson manifold [2, Def. 2.1] (M, π ) defines a Lie algebroid structure on T ∗ M ⊕ g, where g is the Lie algebra of the Lie group acting on M. The leaves of this Lie algebroid coincide with the leaves of the “quasi-Hamiltonian foliation’’ of [2, Sec. 9] in the Hamiltonian case, though, in our framework, we make no assumption about the existence of group-valued moment maps. In Section 3, we study Hamiltonian actions in the context of Dirac geometry at the infinitesimal level. We observe that Dirac realizations, like Poisson maps, are always associated with Lie algebroid actions. (This is, in fact, the guiding principle in our definition of Dirac realizations.) After discussing how classical notions of infinitesimal Hamiltonian actions fit into this framework, we prove the main result of the section: Dirac realizations of Cartan–Dirac structures on Lie groups [6, 28] are equivalent to quasi-Poisson g-manifolds carrying group-valued moment maps. This equivalence involves an “inversion’’procedure relating twisted Dirac structures and quasi-Poisson bivectors, revealing that these two objects are in a certain sense “mirror’’ to one another. The main ingredients in this discussion are the Lie algebroids of Section 2 and the bundle maps which appear in [6] as infinitesimal versions of multiplicative 2forms. This result explains, in particular, the relationship between Cartan–Dirac and quasi-Poisson structures on Lie groups; on the other hand, it recovers the correspondence proved in [2, Thm. 10.3] between “nondegenerate’’ Hamiltonian quasi-Poisson

Dirac structures, momentum maps, and quasi-Poisson manifolds

3

manifolds (i.e., those for which the Lie algebroids of Section 2 are transitive) and quasi-Hamiltonian spaces [3]. In Section 4, we study moment maps in Dirac geometry from a global point of view. We show that complete Dirac realizations “integrate’’to presymplectic groupoid actions, which are natural extensions of those studied in [33]. As our main example, we show that the “integration’’ of Dirac realizations of Cartan–Dirac structures on Lie groups results in Hamiltonian quasi-Poisson G-manifolds. Finally, we show that the natural reduction procedure in the setting of Dirac geometry encompasses various classical reduction theorems [21, 24, 25] as well as their “quasi’’ counterparts [2, 3, 33]. We remark, following an observation of E. Meinrenken, that the results concerning quasi-Poisson manifolds in this paper only require the Lie algebras to be quadratic, in contrast with some of the constructions in [2], in which the positivity of the bilinear forms plays a key role. (In particular, our results hold for quasi-Poisson G-manifolds when G is a noncompact semisimple Lie group.) Most of our constructions can be carried out in the more general setting of [1], but this will be discussed in a separate paper. A work which gave initial motivation and is closely related to the present paper is that of Xu [33], in which a Morita theory of quasi-symplectic groupoids is developed in order to compare “moment map theories.’’ Our results show that twisted Dirac structures complement Xu’s picture in two ways: on the one hand, by providing the infinitesimal framework for Morita equivalence; on the other hand, by leading to more general “modules’’ (i.e., Hamiltonian spaces). It is a pleasure to dedicate this paper to Alan Weinstein, whose work and insightful ideas have been an unlimited source of inspiration to us. Notation. We use the following conventions for bundle maps: if π is a bivector field on M, then π : T ∗ M → T M, α → π(α, ·); if ω is a 2-form, then ω : T M → T ∗ M, X → ω(X, ·). The space of k-multivector fields on M is denoted by X k (M). On a Lie group G, with Lie algebra g, (·, ·)g will denote a bi-invariant nondegenerate quadratic form; we write φ G for the associated Cartan 3-form, and χG ∈ 3 g for the dual trivector. The Lie algebra g is identified with right-invariant vector fields on G.

2 Lie algebroids, bivector fields, and Poisson geometry 2.1 Lie algebroids A Lie algebroid over a manifold M is a vector bundle A → M together with a Lie algebra bracket [·, ·] on the space of sections (A), and a bundle map ρ : A → T M, called the anchor, satisfying the Leibniz identity [ξ, f ξ ] = f [ξ, ξ ] + Lρ(ξ ) (f )ξ

for ξ, ξ ∈ (A)

and

f ∈ C ∞ (M). (2.1)

Whenever there is no risk of confusion, we will write Lρ(ξ ) simply as Lξ .

4


If M is a point, then a Lie algebroid over M is a Lie algebra in the usual sense. An important feature of Lie algebroids A → M is that the image of the anchor, ρ(A) ⊆ T M, defines a generalized integrable distribution, determining a singular foliation of M. The leaves of this foliation are the orbits of the Lie algebroid. The following example plays a key role in the study of Hamiltonian actions and moment maps. Example 2.1 (transformation Lie algebroids). Consider an infinitesimal action of a Lie algebra g on a manifold M, given by a Lie algebra homomorphism ρ¯ : g → X (M). The transformation Lie algebroid associated with this action is the trivial vector bundle M × g, with anchor (x, v) → ρ(x, v) := ρ(v)(x) ¯ and Lie bracket on (M × g) = C ∞ (M, g) defined by [u, v](x) := [u(x), v(x)]g + (ρ(u(x)) ¯ · v)(x) − (ρ(v(x)) ¯ · u)(x).

(2.2)

We often denote a transformation Lie algebroid by g M. Note that [·, ·] is uniquely determined by the condition that it coincides with [·, ·]g on constant functions and the Leibniz identity. The orbits of g M are the g-orbits on M. The remainder of this section is devoted to examples of Lie algebroids closely related to Poisson manifolds. 2.2 Bivector fields and Poisson structures If (M, π ) is a Poisson manifold, then T ∗ M carries a Lie algebroid structure with anchor π : T ∗ M → T M, β(π (α)) = π(α, β), (2.3) and bracket [α, β] = Lπ (α) (β) − Lπ (β) (α) − dπ(α, β),

(2.4)

uniquely characterized by [df, dg] = d{f, g} and the Leibniz identity (2.1). Here, as usual, {f, g} = π(df, dg) is the Poisson bracket on C ∞ (M). In this case, the orbits of T ∗ M are the symplectic leaves of M, i.e., the integral manifolds of the distribution defined by the Hamiltonian vector fields Xf = π (df ). Example 2.2 (Lie–Poisson structures). Let (g, [·, ·]) be a Lie algebra, and consider g∗ equipped with the associated Lie–Poisson structure {f, g}(µ) := µ, [df (µ), dg(µ)], µ ∈ g∗ .

(2.5)

Under the identification T ∗ g∗ ∼ = g∗ ×g, one can see that the Lie algebroid structure on ∗ ∗ T g induced by (2.5) is that of a transformation Lie algebroid g g∗ (see Example 2.1) and a direct computation reveals that the action in question is the coadjoint action.


5

If π ∈ X 2 (M) is an arbitrary bivector field, let us consider π , [·, ·], {·, ·} and Xf as defined by the previous formulas, and let χπ ∈ X 3 (M) be the trivector field defined by χπ := [π, π], (2.6) i.e., χπ satisfies 1 χπ (df, dg, dh) = {f, {g, h}} + {g, {h, f }} + {h, {f, g}} = {f, {g, h}} + c.p., 2 where we use c.p. to denote cyclic permutations. Lemma 2.3. For any bivector field π on M, one has 1 π ([α, β]) = [π (α), π (β)] − iα∧β (χπ ), 2 1 [α, [β, γ ]] + c.p. = (Liα∧β (χπ ) (γ ) + c.p.) − d(χπ (α, β, γ )), 2

(2.7) (2.8)

for α, β, γ ∈ 1 (M). As a result, the following are equivalent: (i) π is a Poisson tensor; (ii) π : 1 (M) → X (M) preserves the brackets; (iii) the bracket [·, ·] on 1 (M) satisfies the Jacobi identity; (iv) (T ∗ M, π , [·, ·]) is a Lie algebroid. Proof. The key remark is that the difference between the left- and right-hand sides of each of (2.7) and (2.8) is C ∞ (M)-multilinear in α, β and γ . So it is enough to prove the identities on exact forms, which is immediate.

Example 2.4 (twisted Poisson manifolds). Consider a closed 3-form φ ∈ 3 (M). A φ-twisted Poisson structure on M [19, 27] consists of a bivector field π ∈ X 2 (M) satisfying 1 [π, π] = π (φ). 2 Here, we abuse notation and write π to denote the map induced by (2.3) on exterior algebras. We know from Lemma 2.3 that the bracket (2.4) induced by π is not preserved by π and does not satisfy the Jacobi identity. However, π ([α, β] + iπ (α)∧π (β) (φ)) = [π (α), π (β)]. Hence, if we define a “twisted’’ version of the bracket (2.4), [α, β]φ := [α, β] + iπ (α)∧π (β) (φ), then π will preserve this new bracket, and [·, ·]φ satisfies the Jacobi identity. As a result, (T ∗ M, π , [·, ·]φ ) is a Lie algebroid. We leave it to the reader to prove a “twisted’’ version of Lemma 2.3.

6


2.3 The Lie algebroid of a quasi-Poisson manifold Let G be a Lie group with Lie algebra g, equipped with a bi-invariant nondegenerate quadratic form (·, ·)g . Let φ G be the bi-invariant Cartan 3-form on G, and let χG ∈ 3 g be its dual trivector. On Lie algebra elements u, v, w ∈ g, we have φ G (u, v, w) = χG (u∨ , v ∨ , w∨ ) =

1 (u, [v, w])g , 2

where u∨ , v ∨ , w∨ are dual to u, v, w via (·, ·)g ; when (·, ·)g is a metric and ea is an orthonormal basis of g, we can write1 χG =

1 (ea , [eb , ec ])g ea ∧ eb ∧ ec . 12

A quasi-Poisson G-manifold [2] consists of a G-manifold M together with a Ginvariant bivector field π satisfying χπ = ρM (χG ),

(2.9)

where ρM : g −→ X (M) is the associated infinitesimal action, and we keep the same notation for the induced maps of exterior algebras. When M is just a g-manifold, we call the corresponding object a quasi-Poisson g-manifold. The two notions are related by the standard procedure of integration of infinitesimal actions; in particular, they coincide if M is compact and G is simply connected. In analogy with ordinary or twisted Poisson manifolds, are quasi-Poisson structures also associated with Lie algebroids? As we now discuss, the answer is yes. Let us consider a more general setup: let M be a g-manifold and let π ∈ X 2 (M) be an arbitrary bivector field. Motivated by [2, Sec. 9], we consider on T ∗ M ⊕ g the “anchor’’ map r : T ∗ M ⊕ g −→ T M, r(α, v) = π (α) + ρM (v),

(2.10)

combining the bivector field and the action. On sections of T ∗ M ⊕ g, we consider the bracket defined by 1 [(α, 0), (β, 0)] = [α, β], iρM∗ (α∧β) (χG ) , (2.11) 2 [(0, v), (0, v )] = (0, [v, v ]), (2.12) [(0, v), (α, 0)] = (LρM (v) (α), 0), (2.13) for all 1-forms α, β ∈ 1 (M) and all v, v ∈ g (thought of as constant sections in C ∞ (M, g)). As in Example 2.1, the definition of the bracket on general elements in (T ∗ M ⊕ g) = 1 (M) ⊕ C ∞ (M, g) is obtained from the Leibniz formula (2.1). With these definitions, we obtain a quasi-Poisson analogue of Lemma 2.3. 1 More generally, with no positivity assumptions on (·, ·) , we can write χ g G = 1 (e , [e , e ]) f ∧ f ∧ f , where f is a basis of g satisfying (f , e ) = δ . a c g a c a a g b b b ab 12

A similar observation holds for (2.25).


7

Theorem 2.5. Let M be a g-manifold equipped with a bivector field π . The following are equivalent: (i) (M, π ) is a quasi-Poisson g-manifold; (ii) r : 1 (M) ⊕ C ∞ (M, g) → X (M) preserves brackets; (iii) the bracket [·, ·] on 1 (M) ⊕ C ∞ (M, g) satisfies the Jacobi identity; (iv) (T ∗ M ⊕ g, r, [·, ·]) is a Lie algebroid. Proof. Note that r preserves the bracket (2.12), since ρM is an action. From the identity (2.7) in Lemma 2.3, it follows that r preserves the bracket of type (2.11) if and only if χπ = ρM (χG ). On the other hand, r preserves the bracket of type (2.13) if and only if π LρM (v) (ξ ) = LρM (v) π (ξ ), which is equivalent to the g-invariance of π. This shows that (i) and (ii) are equivalent. Let us prove that (i) implies (iii); from the proof, the converse will be clear. Assuming (i), we must show that [·, ·] on 1 (M) ⊕ C ∞ (M, g) satisfies the Jacobi identity. On elements of type (0, v), this reduces to the Jacobi identity for g (or, alternatively, for g M). On elements (0, v), (0, w) and (α, 0), the Jacobi identity of [·, ·] reduces to the fact that ρM is an action. Computing the “jacobiator’’ for elements of type (0, v), (α, 0), (β, 0), we see that the first component is [LρM (v) (α), β] + [α, LρM (v) (β)] − LρM (v) ([α, β]).

(2.14)

Using the Leibniz identity, we see that the C ∞ (M)-linearity of (2.14) with respect to β is equivalent to π Lρ(v) (β) = Lρ(v) π (β), i.e., to the g-invariance of π . Hence, if π is invariant, (2.14) is C ∞ (M)-linear on α and β, and then one can check that it is zero by looking at the particular case when α and β are exact. The second component of the jacobiator of (0, v), (α, 0), (β, 0) can be computed similarly. To complete the proof that (i) implies (iii), we must deal with the Jacobi identity for elements of type (α, 0), (β, 0), (γ , 0). To this end, we first need to find the expression for the bracket between elements of type (0, v) ˜ and (α, 0), with v˜ ∈ C ∞ (M, g) not 1 necessarily constant: pairing d v˜ ∈ (M; g) with an element µ ∈ C ∞ (M, g∗ ) gives us a 1-form on M, denoted by Av˜ (µ), satisfying the following two properties: Af v˜ (µ) = f Av˜ (µ) + µ(v)df, ˜ and

Av˜ (f µ) = f Av˜ (µ),

for f ∈ C ∞ (M). We claim that ∗ [(0, v), ˜ (α, 0)] = (LρM (v) ˜ ˜ (α) − Av˜ (ρM (α)), −Lπ (α) (v)).

(2.15)

To see this, note that (2.15) holds when v˜ is constant, and the difference between the left- and right-hand sides is C ∞ (M)-linear in v. ˜ We remark that Aiµ∧µ (χG ) (µ ) + c.p. = 2d(χG (µ, µ , µ )).

(2.16)

Again, it is easy to check this identity when µ, µ and µ are constant, so (2.16) follows from C ∞ (M)-linearity. Also, denoting χM := ρM (χG ), a direct computation shows that

8


ρM (iρM∗ (α∧β) (χG )) = iα∧β (χM ). We now turn to the computation of the jacobiator of the elements (α, 0), (β, 0) and (γ , 0), that we denote by Jac(α, β, γ ). For the first component of Jac(α, β, γ ), we obtain 1 1 ∗ (γ ))+c.p.). (2.17) ([α, [β, γ ]]+c.p.)− (Liα∧β (χM ) (γ )+c.p.)+ (Aiα∧β (χM ) (ρM 2 2 Combining the second identity of Lemma 2.3 with (2.16), we get that (2.17) equals d((ρM (χG ) − χπ )(α, β, γ )), which vanishes by the condition χπ = ρM (χG ). So we are left with proving that the second component of Jac(α, β, γ ) vanishes, which amounts to showing that iρM∗ ([α,β]∧γ ) (χG ) + c.p. = Lπ (γ ) iρM∗ (α∧β) (χG ) + c.p..

(2.18)

In order to do that, consider the operators iρM∗ ([α,β]) and Lπ (α) iρM∗ (β) − Lπ (β) iρM∗ (α) acting on C ∞ (M, g), for α, β ∈ 1 (M). Claim 2.6. On g, seen as constant functions in C ∞ (M, g), we have iρM∗ ([α,β]) = Lπ (α) iρM∗ (β) − Lπ (β) iρM∗ (α) .

(2.19)

Proof. Both operators are derivations of degree −1 on g, hence it suffices to show (2.19) for elements v ∈ g. As we now check, this follows from the definition of the bracket induced by π and the invariance of π: on the one hand, iρM∗ ([α,β]) (v) = [α, β](ρM (v)) = iρM (v) Lπ (α) (β) − iρM (v) Lπ (β) (α) − iρM (v) dπ(α, β).

(2.20)

Using that i[X,Y ] = LX iY − iY LX for vector fields X, Y , we have iρM (v) Lπ (α) (β) = Lπ (α) (β(ρM (v))) − β([π (α), ρM (v)]) = Lπ (α) iρM∗ (β) (v) − π(LρM (v) (α), β),

(2.21)

where the last equality follows from the g-invariance of π . Using the identity (2.21) (and its analogue for α and β interchanged) in (2.20), (2.19) follows.

Using the claim, we see that iρM∗ ([α,β]∧γ ) + c.p. = iρM∗ (γ ) iρM∗ ([α,β]) + c.p. = (iρM∗ (γ ) Lπ (α) iρM∗ (β) − iρM∗ (γ ) Lπ (β) iρM∗ (α) ) + c.p., (2.22) when restricted to constant elements in C ∞ (M, g) . On the other hand, it follows from (2.19) that, on g, we can write iρM∗ ([α,β]) = [Lπ (α) , iρM∗ (β) ] − [Lπ (β) , iρM∗ (α) ]

(2.23)


9

since the Lie derivatives are zero on constant functions. But both sides of (2.23) are C ∞ (M)-linear, so this equality is valid for all C ∞ (M, g). So we can write iρM∗ ([α,β]∧γ ) + c.p. = −iρM∗ ([α,β]) iρM∗ (γ ) + c.p. = −([Lπ (α) , iρM∗ (β) ] − [Lπ (β) , iρM∗ (α) ])iρM∗ (γ ) + c.p., from which we deduce that iρM∗ ([α,β]∧γ ) + c.p. = 2(Lπ (α) iρM∗ (β∧γ ) + c.p.) − (iρM∗ (γ ) Lπ (α) iρM∗ (β) − iρM∗ (β) Lπ (α) iρM∗ (γ ) + c.p.). On constant functions, we can use (2.22) to conclude that (iρM∗ ([α,β]∧γ ) + c.p.) = 2(Lπ (α) iρM∗ (β∧γ ) + c.p.) − (iρM∗ ([α,β]∧γ ) + c.p.), i.e., iρM∗ ([α,β]∧γ ) + c.p. = Lπ (α) iρM∗ (β∧γ ) . Evaluating this identity at χG proves (2.18), showing that (i) implies (iii). Looking back at the proof, one can check that the same formulas show the converse, so that (i) and (iii) are equivalent. Since (iii) and the Leibniz identity for [·, ·] are together equivalent to (iv), it follows that (i)–(iv) are equivalent to each other.

Corollary 2.7. If (M, π ) is a quasi-Poisson g-manifold, then the generalized distribution π (α) + ρM (v) ⊆ T M, for α ∈ T ∗ M, v ∈ g, is integrable. This result shows that the singular distribution discussed in [2, Thm. 9.2] in the context of Hamiltonian quasi-Poisson manifolds is integrable even without the presence of a moment map (and without the positivity of (·, ·)g ). As in the case of ordinary Poisson manifolds, we call a quasi-Poisson manifold nondegenerate if its associated Lie algebroid is transitive (i.e., its anchor map is onto). Example 2.8 (quasi-Poisson structures on Lie groups). Let G be a Lie group with Lie algebra g, which we assume to be equipped with an invariant nondegenerate quadratic form (·, ·)g . We consider G acting on itself by conjugation. As shown in [2, Sec. 3], the bivector field πG , defined on left invariant 1-forms by πG (dlg∗−1 (µ), dlg∗−1 (ν)) :=

1 ((Ad g −1 − Ad g )(µ∨ ), ν ∨ )g , 2

(2.24)

where lg denotes left multiplication by g ∈ G, µ, ν ∈ g∗ , and µ∨ is the element in g dual to µ via (·, ·)g , makes G into a quasi-Poisson G-manifold. If (·, ·)g is a metric, then we can write 1 l πG = (2.25) ea ∧ ear , 2 where ea is an orthonormal basis of g and ear (respectively, eal ) are the corresponding right (respectively, left) translations.

10


In this example, the image of πG is tangent to the G-orbits, so the leaves of the corresponding foliation are the conjugacy classes. The formula for the Lie algebroid bracket on T ∗ G ⊕ g bears close resemblance with the one for the bracket in the “double’’ of the Lie quasi-bialgebra of G, as in [4]. We will discuss this connection in a separate work.

3 Moment maps in Dirac geometry: The infinitesimal picture 3.1 Dirac manifolds Let φ be a closed 3-form on a manifold M. A φ-twisted Dirac structure on M [28] is a subbundle L ⊂ E = T M ⊕ T ∗ M satisfying the following two conditions: 1. L is maximal isotropic with respect to the symmetric pairing ·, ·+ : (E) × (E) → C ∞ (M), (X, α), (Y, β)+ := β(X) + α(Y );

(3.1)

2. The space of sections (L) is closed under the bracket [[·, ·]]φ : (E) × (E) → (E), [[(X, α), (Y, β)]]φ := ([X, Y ], LX β − iY dα + iX∧Y φ). (3.2) Since the pairing (3.1) has zero signature, condition 1 is equivalent to requiring that L has rank equal to dim(M) and that ·, ·+ |L = 0. The bracket (3.2) is the φ-twisted Courant bracket considered in [28]. When φ = 0, this bracket is a nonskew-symmetric version of Courant’s original bracket introduced in [12]. Twisted Dirac structures are always associated with Lie algebroids. Indeed, the restriction of the Courant bracket [[·, ·]]φ to a Dirac subbundle L ⊂ T M ⊕ T ∗ M defines a Lie algebra bracket on the space of sections (L), making L → M into a Lie algebroid with anchor ρ = pr 1 |L : L → T M, where pr 1 is the first projection. The orbits of this algebroid are also called the leaves of L. Example 3.1 (twisted Poisson structures). If π is a bivector field on M, then Lπ := graph(π ) ⊂ T M ⊕ T ∗ M satisfies condition 1, and Lπ is a φ-twisted Dirac structure if and only if π is a φ-twisted Poisson structure in the sense of Example 2.4. In this case, the second projection pr 2 |L : L → T ∗ M establishes an isomorphism of Lie algebroids, where T ∗ M is equipped with the Lie algebroid structure described in Example 2.4. Setting φ = 0, we obtain a one-toone correspondence between ordinary Poisson structures on M and Dirac structures satisfying the extra condition L ∩ T M = {0}.


11

Example 3.2 (twisted presymplectic forms). Similarly, the graph associated with a 2-form ω ∈ 2 (M), Lω = graph(ω ), is a φ-twisted Dirac structure if and only if dω + φ = 0, and we refer to ω as a φ-twisted presymplectic form. In this case, setting φ = 0, we have an identification of closed 2-forms on M with Dirac structures satisfying L ∩ T ∗ M = {0}. In general, the leaves of a φ-twisted Dirac structure L carry twisted presymplectic forms defined as follows: at each x ∈ M, we define a skew symmetric bilinear form θx on ρ(L)x = pr 1 (L)x by θx (X1 , X2 ) = α(X2 ),

(3.3)

where α is any element in Tx∗ M satisfying (X1 , α) ∈ Lx . The fact that L is maximal isotropic with respect to (3.1) guarantees that (3.3) is independent of the choice of α, and these forms fit together into a smooth leafwise 2-form θ. Using that (L) is closed with respect to (3.2), one can show that on each leaf ι : O → M, the 2-form θ satisfies dθ + ι∗ φ = 0. At each point x ∈ M, the kernel of θ coincides with Lx ∩ Tx M, which shows that the leafwise presymplectic forms are nondegenerate if and only if L comes from a φ-twisted Poisson structure. We will denote the distribution L ∩ T M on M by ker(L). Since Dirac structures are always associated with Lie algebroids, it is natural to consider how to obtain Dirac structures from them. The following is a useful construction, see [6]: for a Lie algebroid A over M with anchor ρ : A −→ T M, we define a φ-IM form of A to be any bundle map2 σ : A −→ T ∗ M satisfying the following properties: (3.4) σ (ξ ), ρ(ξ ) = −σ (ξ ), ρ(ξ ); σ ([ξ, ξ ]) = Lξ (σ (ξ )) − Lξ (σ (ξ )) + dσ (ξ ), ρ(ξ ) + iρ(ξ )∧ρ(ξ ) (φ), (3.5) for ξ, ξ ∈ (A) (here ·, · denotes the usual pairing between a vector space and its dual). Let Lσ ⊂ T M ⊕ T ∗ M be the image of the map (ρ, σ ) : A −→ T M ⊕ T ∗ M. Then the following is immediate. Lemma 3.3. If σ is a φ-IM form of A and rank(Lσ ) = dim(M), then Lσ is a φ-twisted Dirac structure on M. Of course, any Dirac structure can be realized as the image of an IM form by taking A = L, viewed as an algebroid with ρ = pr 1 |L, and σ = pr 2 |L. The following is a key example. 2 These bundle maps are infinitesimal versions of multiplicative 2-forms on groupoids; see

[6]; the terminology “IM’’ stands for “infinitesimal multiplicative.’’

12


Example 3.4 (Cartan–Dirac structures on Lie groups). Cartan–Dirac structures on Lie groups play a role in Dirac geometry analogous to the one played by Lie–Poisson structures (Example 2.2) in Poisson geometry. Just as Lie–Poisson structures on the dual of Lie algebras are completely determined by the Kostant–Kirillov–Souriau (KKS) symplectic forms along coadjoint orbits, Cartan–Dirac structures on Lie groups “assemble’’ certain 2-forms defined on conjugacy classes defined as follows. Let G be a Lie group with Lie algebra g, and let (·, ·)g be a bi-invariant nondegenerate quadratic form, which we use to identify T G and T ∗ G. For v ∈ g, let vG = vr −vl be the infinitesimal generator of the action of G on itself by conjugation. On each conjugacy class, we define ι : C → G, a 2-form θ by 1 (Ad g − Ad g −1 )u, v , g ∈ C. θg (uG , vG ) := (3.6) 2 g Direct computations show that dθ − ι∗ φ G = 0, where φ G is the bi-invariant Cartan 3-form on G, and that θg is nondegenerate at a point g if and only if (Ad g + 1) is invertible. The 2-forms (3.6) appear in [17] in the study of symplectic structures of moduli spaces. Since these 2-forms are not symplectic, but twisted presymplectic, they should correspond to a −φ G -twisted Dirac structure LG on G rather than a Poisson structure. A simple computation shows that 1 vr − vl , (vr + vl ) , v ∈ g ⊂ T G ⊕ T G. (3.7) LG = 2 (Recall that we are identifying T G with T ∗ G via (·, ·)g .) We call LG the Cartan– Dirac structure on G associated with (·, ·)g [28, 6]. Note that ρ(v) = vr − vl is the anchor of the action Lie algebroid (Example 2.1) g G with respect to the action by conjugation, and the map σ : G × g −→ T G, σ (v) =

1 (vr + vl ) 2

(3.8)

satisfies the conditions of Lemma 3.3. So σ is a −φ G -IM form of g G, and the Cartan–Dirac structure LG arises as the image of (ρ, σ ). In this case, (ρ, σ ) actually establishes an isomorphism between g G and LG . (Note the analogy with Example 2.2, which shows that Lie algebroids of Lie–Poisson structures are isomorphic to the action Lie of algebroids for the coadjoint action!) Let us finally recall an important operation involving Dirac structures: if L is a φ-twisted Dirac structure on M and B ∈ 2 (M), then τB (L) := {(X, α + B (X)) | (X, α) ∈ L}

(3.9)

defines a (φ − dB)-twisted Dirac structure on M [28]. The operation τB is called a gauge transformation associated with B, and it has the effect of modifying L by adding the pullback of B to the presymplectic form on each leaf.


13

3.2 Dirac maps Since Dirac structures generalize both Poisson and presymplectic structures, we have two possible definitions of Dirac maps; see [7]. Let (M, LM ) and (N, LN ) be twisted Dirac manifolds.Asmooth map f : N → M is a forward Dirac map, or f-Dirac in short, if LN and LM are related as follows: LM = {(df (Y ), α) | Y ∈ T N, α ∈ T ∗ M and (Y, df ∗ (α)) ∈ LN }.

(3.10)

If LM and LN are associated with twisted Poisson structures, then an f-Dirac map is equivalent to a Poisson map. The terminology “forward’’ is due to the fact that, at each point, (3.10) extends the usual notion of “push-forward’’ of a linear bivector. For this reason, we may write LM = f∗ LN instead of (3.10), in analogy with the notation for “f -related’’ bivector fields on a manifold. Similarly, f : N → M is a backward Dirac map, or simply b-Dirac, if LN = {(Y, df ∗ α) | Y ∈ T N, α ∈ T ∗ M and (df (Y ), α) ∈ LM }.

(3.11)

If LM and LN are associated with twisted presymplectic structures ωM and ωN , then a b-Dirac map is just a map satisfying f ∗ ωM = ωN . As before, we will write LN = f ∗ LM to denote that f is a b-Dirac map. Note that f ∗ LM is always a well-defined, though not necessarily smooth, subbundle of T N, in contrast with f∗ LN , which may not be well defined at all. In fact, f ∗ LM defines a Dirac structure on N provided it is smooth, which is the case, e.g., when f is a submersion. However, as illustrated in the next example, f ∗ LM may define a Dirac structure even when f is not a submersion. Example 3.5 (inclusion of presymplectic leaves). Let L be a twisted Dirac structure on M, and consider a presymplectic leaf O, equipped with Dirac structure Lθ associated with the twisted presymplectic form θ. Denoting by ι : O → M the inclusion map, it follows from the definition of θ that Lθ = {(X, iX θ ) | X ∈ T O} = {(X, (dι)∗ α) | (dι(X), α) ∈ L} = ι∗ L.

(3.12)

So ι : (O, Lθ ) → (M, L) is a b-Dirac map. On the other hand, at each point of M, we have ι∗ Lθ = {(dι(X), α) | (X, (dι)∗ α) ∈ Lθ }. By the second equality in (3.12), it follows that ι∗ Lθ ⊆ L, but since they have the same dimension, we get ι∗ Lθ = L, (3.13) so ι is f-Dirac as well.

14


Note that the fact that the inclusion of presymplectic leaves into a Dirac manifold is an f-Dirac map is a direct generalization of the fact that the inclusion of symplectic leaves into a Poisson manifold is a Poisson map. As a simple consequence, we have the following. Corollary 3.6. Let (N, LN ) and (M, LM ) be twisted Dirac manifolds. A map J : N → M is f-Dirac if and only if its restriction to each presymplectic leaf of N is f-Dirac. We remark that Example 3.5 is very special in that the inclusion map of presymplectic leaves is both forward and backward Dirac (see also Remark 4.12). In general, f-Dirac maps need not be b-Dirac, or the other way around. 3.3 Poisson maps as infinitesimal Hamiltonian actions The usual notion of Lie algebra action can be extended to the realm of Lie algebroids, the main difference being that algebroids, rather than acting on manifolds, act on maps from manifolds into their base [18]: An action of a Lie algebroid A → M on a map J : N → M consists of a Lie algebra homomorphism ρN : (A) → X (N ) satisfying dJ ◦ ρN (ξ ) = ρ(ξ ), for all ξ ∈ (A), (3.14) and such that, for f ∈ C ∞ (M) and ξ ∈ (A), ρN (f ξ ) = J ∗ fρN (ξ ) (i.e., the induced map (J ∗ A) → X (N ) comes from a vector bundle morphism J ∗ A → T N, where J ∗ A = A ×M N is the pullback of the vector bundle A by J ). Example 3.7 (actions of transformations Lie algebroids). Consider an infinitesimal action ρ of g on a manifold M. Then an action ρN of the transformation Lie algebroid A = g M on a map J : N → M is equivalent to an infinitesimal action ρN of g on N for which J is g-equivariant. Indeed, ρN and ρN are related by the formula ρN (v)y = ρN (v(J (y)))y , where v ∈ C ∞ (M, g), y ∈ N,

(3.15)

and the g-equivariance of J corresponds to (3.14). In Poisson geometry, Poisson maps are always associated with Lie algebroid actions: If (Q, πQ ) and (P , πP ) are Poisson manifolds, then any Poisson map J : Q → P induces a Lie algebroid action of T ∗ P on Q by

1 (P ) −→ X (Q),

α → πQ (J ∗ α).

(3.16)

When the target P is the dual of a Lie algebra, we recover a familiar example. Example 3.8 (infinitesimal Hamiltonian actions). Consider g∗ equipped with its Lie– Poisson structure. As remarked in Example 2.2, the Lie algebroid structure on T ∗ g∗ induced by (2.5) is that of a transformation Lie algebroid g g∗ with respect to the coadjoint action. If J : Q → g∗ is a Poisson map, then it induces an action of T ∗ g∗ via (3.16), which, by Example 3.7, is equivalent to an ordinary g-action on Q for which J is equivariant. A simple computation shows that the g-action arising in this way is just a Hamiltonian action in the usual sense, making Q into a Hamiltonian Poisson g-manifold having J as a momentum map.


15

Recall that a Poisson map J : Q → P is called a symplectic realization if Q is symplectic. The following is an immediate consequence. Proposition 3.9. There is a one-to-one correspondence between Poisson maps into g∗ and Hamiltonian Poisson g-manifolds, and this correspondence restricts to a one-to-one correspondence between symplectic realizations of g∗ and Hamiltonian symplectic g-manifolds. Remark 3.10. An analogue of Proposition 3.9 holds more generally in the context of Poisson–Lie groups [20, 22]. Let (G, π) be a simply connected Poisson–Lie group, and let G∗ be its dual. The Lie algebroid structure on T ∗ G∗ ∼ = G∗ × g induced from the dual Poisson structure is a transformation Lie algebroid, now associated with the infinitesimal dressing action of g on G∗ . For a Poisson map J : Q → G∗ , the general Lie algebroid action described by (3.16) reduces to a Poisson g-action for which J is an equivariant momentum map in the sense of Lu [21]. In order to extend this discussion to Dirac geometry, let us consider LπP = graph(πP ), the associated Dirac structure on (P , πP ). Using the Lie algebroid isomorphism T ∗ P ∼ = LπP , we can rewrite the infinitesimal action (3.16) as (LπP ) → X (Q), (X, α) → Y,

(3.17)

where Y ∈ X (Q) is uniquely determined by the condition (Y, J ∗ α) ∈ LπQ . Also note that Y is related to X by dJ (Y ) = X, since J is a Poisson map. The question of whether this procedure can be carried out for f-Dirac maps leads us to the notion of Dirac realization. 3.4 Dirac realizations If (N, LN ) and (M, LM ) are twisted Dirac manifolds, then, by definition, a smooth J : N → M is an f-Dirac map if and only if, given (X, α) ∈ (LM )J (y) , there exists a Y ∈ Ty N with the property that (Y, dJ ∗ α) ∈ (LN )y and X = (dJ )y (Y ).

(3.18)

It is natural to try to define an action of LM on N as in the case of Poisson maps, see (3.17), except that (3.18) does not determine Y uniquely in general. In fact, this is the case if and only if the following extra “nondegeneracy’’ condition holds: ker(dJ ) ∩ ker(LN ) = {0}.

(3.19)

A similar argument as in [6, Section 7.1] shows that (3.19) is equivalent to J : ker(LN ) → ker(LM ) being an isomorphism. Definition 3.11. A Dirac realization of a φ-twisted Dirac manifold (M, LM ) is an f-Dirac map J : (N, LN ) → (M, LM ), where LN is a J ∗ φ-twisted Dirac structure on N, satisfying (3.19).

16


As a consequence of Definition 3.11, we have the following. Corollary 3.12. Let J : N → M be a Dirac realization. Then the map (LM ) → X (N), (X, α) → Y , where Y is determined by the conditions in (3.18), is a Lie algebroid action. Dirac realizations J : N → M for which N is presymplectic were studied in [6, Sec. 7.1] under the name of presymplectic realizations. As a result of Corollary 3.6, we have the following. Corollary 3.13. A map J : N → M is a Dirac realization if and only if its restriction to each presymplectic leaf of N is a presymplectic realization. Similar to Poisson geometry, the connection between Dirac realizations and “Hamiltonian actions’’ is established by a suitable choice of “target’’ M. Following the analogy between Lie–Poisson structures and Cartan–Dirac structures, it is natural to study the “Hamiltonian spaces’’ associated with Dirac realizations of Cartan– Dirac structures. The particular case of presymplectic realizations is discussed in [6, Sec. 7.2]. Example 3.14 (presymplectic realizations of Cartan–Dirac structures). Let G be a Lie group with Lie algebra g, equipped with a bi-invariant nondegenerate quadratic form (·, ·)g . Let LG be the associated Cartan–Dirac structure on G. If (M, ωM ) is a twisted presymplectic manifold, then the conditions for J : M → G being a presymplectic realization can be expressed as follows: 1. ωM is g-invariant and satisfies dωM = J ∗ φ G ; 2. at each x ∈ M, Ker(ωM )x = {(ρM )x (v) : v ∈ Ker(Ad J (p) + 1)}; 3. the map J satisfies the moment map condition ω ρM = J ∗ σ.

(3.20)

The invariance of ωM in 1 is with respect to the g-action ρM induced by J (recall that LG ∼ = g G, see Example 3.4, so an LG -action defines an ordinary g-action), for which J is equivariant; in 3, σ is the IM-form of the Cartan–Dirac structure (3.8), σ : g −→ T ∗ G,

σ (v) =

1 (vr + vl )∨ , 2

(3.21)

where v −→ v ∨ denotes the isomorphism T G −→ T ∗ G induced by the quadratic form. The “relative closedness’’ of ωM in 1 expresses that the associated Dirac structure is −J ∗ φ G -twisted, while condition 2 is the “nondegeneracy’’condition (3.19) applied to this particular case; finally, condition 3 follows from J being an f-Dirac map. Conditions 1, 2, and 3 are exactly the defining axioms of a quasi-Hamiltonian gspace, in the sense of [3], for which J is the group-valued moment map. Conversely, any group-valued moment map of a quasi-Hamiltonian g-space is a presymplectic realization of (G, LG ).


17

We summarize Example 3.14 in the next result, analogous to Proposition 3.9; see [6, Thm. 7.6]. Theorem 3.15. There is a one-to-one correspondence between presymplectic realizations of G endowed with the Cartan–Dirac structure, and quasi-Hamiltonian gmanifolds. Combining Corollary 3.13 with Theorem 3.15, we conclude that general Dirac realizations of Cartan–Dirac structures must be “foliated’’ by quasi-Hamiltonian gmanifolds. Since Hamiltonian quasi-Poisson manifolds, in the sense of [2], also have this property [2, Sec. 10], we are led to investigate the relationship between these objects. 3.5 Dirac realizations and Hamiltonian quasi-Poisson g-manifolds 3.5.1 The equivalence theorem For a quasi-Poisson g-manifold (M, π), a momentum map is a g-equivariant map J : M −→ G (with respect to the infinitesimal action by conjugation on G) satisfying the condition [2, Lem. 2.3] π J ∗ = ρM σ ∨ , (3.22) where

1 (dr −1 (ξg∨ ) + dlg −1 (ξg∨ )) (3.23) 2 g is the adjoint of σ (3.21) with respect to the form (·, ·)g , and ρM : g → T M is the gaction. Here lg and rg denote the left and right translations by g, respectively, and, as in Example 3.14, the symbol ∨ on elements of T ∗ G is used to denote the corresponding element in T G via the identification induced by (·, ·)g (and vice versa). The following is our main result in this section. σ ∨ : T ∗ G −→ g,

σ ∨ (ξg ) =

Theorem 3.16. There is a one-to-one correspondence between Dirac realizations of G, endowed with the Cartan–Dirac structure, and Hamiltonian quasi-Poisson gmanifolds. Before proving Theorem 3.16, let us collect some useful formulas relating the maps σ , σ ∨ , ρ : g → T G, ρ(v) = vr − vl , and, for symmetry, the dual of ρ with respect to (·, ·)g , ρ ∨ : T G −→ g,

ρ ∨ (Vg ) = drg −1 (Vg ) − dlg −1 (Vg ).

(3.24)

The following lemma follows from a straightforward computation. Lemma 3.17. The following formulas hold true: 4σ ∨ σ + ρ ∨ ρ = 4Id g , 4σ σ ∨ + (ρρ ∨ )∗ = 4Id T ∗ G ,

(3.25) (3.26)

18


σ ∗ ρ = −ρ ∗ σ, σρ ∨ = −(ρ ∨ )∗ σ ∗ , ∨

∨ ∗

∨

∨ ∗

ρ (σ ) = −σ (ρ ) , ρσ ∨ = −(ρσ ∨ ).∗

(3.27) (3.28) (3.29) (3.30)

Motivated by the equivalence between quasi-Hamiltonian manifolds and nondegenerate Hamiltonian quasi-Poisson manifolds [2, Thm. 10.3], which will also follow from Theorem 3.16, it is natural to combine the two moment map conditions (3.20) and (3.22). By applying π to (3.20) and using (3.22), we obtain, in particular, the relation ρM σ ∨ σ = π ω ρM . This suggests the importance of writing ρM σ ∨ σ as the composition of some operator C : T M → T M with ρM in general. Using (3.25) and the equivariance of J , written as ρ = dJ ◦ ρM , it is easy to find an expression for C (which already appears in [2, Lem. 10.2]). Lemma 3.18. For any manifold M equipped with an infinitesimal action ρM : g −→ T M, and any g-equivariant map J : M −→ G, the operator 1 C = 1 − ρM ρ ∨ (dJ ) : T M −→ T M 4 and its dual C ∗ : T ∗ M −→ T ∗ M satisfy the formulas ρM σ ∨ σ = CρM , and J ∗ σ σ ∨ = C ∗ J ∗ .

(3.31)

Theorem 3.16 follows from the next two propositions, each one describing explicitly one direction of the asserted one-to-one correspondence. Proposition 3.19. Let M be a quasi-Poisson g-manifold, and let A = T ∗ M ⊕ g be its associated Lie algebroid, with anchor r. Then any moment map J : M −→ G induces a −J ∗ φ G -IM form of A by s : A −→ T ∗ M,

s(α, v) = C ∗ (α) + J ∗ σ (v),

(3.32)

so that the image L of the map (r, s) : A −→ T M ⊕ T ∗ M is a −J ∗ φ G -twisted Dirac structure on M, and J : (M, L) −→ (G, LG ) is a Dirac realization of the Cartan–Dirac structure on G. This proposition also suggests the converse construction. Proposition 3.20. Let J : (M, L) −→ (G, LG ) be a Dirac realization of the Cartan– Dirac structure on G. Then (i) for any v ∈ g there is an unique vector V ∈ T M satisfying dJ (V ) = ρ(v) and (V , J ∗ σ (v)) ∈ L;

(3.33)


19

(ii) for any α ∈ T ∗ M, there is an unique vector X ∈ T M satisfying dJ (X) = −(ρM σ ∨ )∗ α, ∗

(X, C (α)) ∈ L.

(3.34) (3.35)

Moreover, v → ρM (v) := V defines a g-action on M, and α → π (α) := X defines a quasi-Poisson tensor π on M so that (M, π) is a Hamiltonian quasi-Poisson gmanifold with moment map J . Note that the g-action defined by (3.33) is the one induced by the infinitesimal LG = g G-action with “moment’’ J : M → G. It is simple to check that the constructions in Propositions 3.19 and 3.20 are inverses to one another. For example, if L is obtained from π as in Proposition 3.19, then L = {(π (α) + ρM (v), C ∗ (α) + J ∗ σ (v)) | α ∈ T ∗ M, v ∈ g}, and it is clear that, given α ∈ T ∗ M, X = π (α) satisfies conditions (3.34) (which is the dual of the moment map condition (3.22)) and (3.35), so Proposition 3.20 constructs π back. Since the proofs of Propositions 3.19 and 3.20 involve long computations, we will postpone them to the next subsection; we will discuss some examples and implications of the results first. Example 3.21 (nondegenerate quasi-Poisson and quasi-Hamiltonian g-manifolds). It is clear from the correspondence constructed in Proposition 3.19 that the singular foliation associated with π, tangent to Im(π ) + Im(ρM ) ⊆ T M, coincides with the singular foliation of the Dirac structure L, tangent to pr 1 (L) ⊆ T M. In other words, the Lie algebroids associated with π and L have the same leaves, so one is transitive if and only if the other one is. Note that, for Dirac structures, pr 1 (L) = T M means exactly that L is defined by a 2-form. As a result, it follows that the correspondence established by Theorem 3.16 restricts to a one-to-one correspondence between nondegenerate Hamiltonian quasi-Poisson manifolds and presymplectic realizations of Cartan–Dirac structures on Lie groups. Combining Example 3.21 with Theorem 3.15, we obtain Corollary 3.22. There is a one-to-one correspondence between (i) nondegenerate quasi-Poisson Hamiltonian g-manifolds, (ii) quasi-Hamiltonian g-manifolds, (iii) presymplectic realizations of G endowed with the Cartan–Dirac structure. Of course, in general, the leaves of a Hamiltonian quasi-Poisson g-manifold are quasi-Hamiltonian g-manifolds, which can now be seen as a particular case of Dirac structures having presymplectic foliations (see also Corollary 3.13). The equivalence of (i) and (ii) can be found in [2]. The next example answers a question posed in [28, Ex. 5.2].

20


Example 3.23 (Cartan–Dirac and quasi-Poisson structures on Lie groups). If G is a Lie group with Lie algebra g equipped with a bi-invariant nondegenerate quadratic form (·, ·)g , then one can regard it as a −φ G -twisted Dirac manifold with respect to the Cartan–Dirac structure LG , or as a Hamiltonian quasi-Poisson g-manifold. In the latter case, we consider G acting on itself by conjugation, the quasi-Poisson tensor is πG , defined in Example 2.8, and the moment map J : G → G is the identity map; see [2, Sec. 3]. We claim that these two structures are “dual’’ to each other in the sense of Theorem 3.16. Indeed, starting with πG and using Proposition 3.19, we see that the corresponding Dirac structure is L = {(πG (α) + ρ(v), C ∗ (α) + σ (v)), | (α, v) ∈ T ∗ M ⊕ g}.

Since LG is the image of (ρ, σ ), it is clear that LG ⊆ L, which implies that LG = L since they have the same dimension. To complete the “duality’’ picture between Dirac realizations of Cartan–Dirac structures and Hamiltonian quasi-Poisson g-manifolds, we note that the correspondence established in Theorem 3.16 preserves maps. If (Mi , πi ) is a Hamiltonian quasi-Poisson g-manifold with moment map Ji : Mi → G, i = 1, 2, then a map f : M1 → M2 is a Hamiltonian quasi-Poisson map if f∗ π1 = π2 , f is g-equivariant, and J2 ◦ f = J1 . Suppose that Li is the Dirac structure on Mi corresponding to πi , i = 1, 2, via Theorem 3.16. Proposition 3.24. A map f : (M1 , π1 ) → (M2 , π2 ) is a Hamiltonian quasi-Poisson map if and only if f : (M1 , L1 ) → (M2 , L2 ) is f-Dirac and commutes with the realization maps, J2 ◦ f = J1 . Proof. Suppose f : M1 → M2 is a Hamiltonian quasi-Poisson map. In order to check that f is f-Dirac, we have to compare L2 , at each point of M2 , with f∗ L1 = {(df (X), β) | (X, df ∗ (β)) ∈ L1 }.

(3.36)

To simplify the notation, we will denote the infinitesimal actions of g on Mi by ρi , and Ci = 1 − (1/4)ρi ρ ∨ dJ , i = 1, 2. Since L2 corresponds to π2 , we have L2 = {(π2 (β) + ρ2 (v), C2∗ (β) + J2∗ σ (v)) | β ∈ T ∗ M2 , v ∈ g}.

Using that df π1 df ∗ = π2 (which is another way of writing f∗ π1 = π2 ) and dfρ1 = ρ2 (which is f g-equivariance), we deduce that

π2 (β) + ρ2 (v) = df (π1 (df ∗ (β)) + ρ1 (v)).

(3.37)

On the other hand, using the g-equivariance of f and J2 ◦ f = J1 , it follows that df C1 = C2 df , and we obtain df ∗ (C2∗ (β) + J2∗ σ (v)) = C1∗ (df ∗ (β)) + J1∗ σ (v).

(3.38)


Since

21

(π1 (df ∗ (β)) + ρ1 (v), C1∗ (df ∗ (β)) + J1∗ σ (v)) ∈ L1 ,

for L1 corresponds to π1 , it follows that, at each point, L2 ⊆ f∗ L1 . But since they have equal dimension, we conclude that L2 = f∗ L1 , so f is forward Dirac. For the converse, suppose that f∗ L1 = L2 and J2 ◦ f = J1 . It is easy to check that, in this case, f is automatically g-equivariant with respect to (3.33). From this, it follows that df C1 = C2 df . In order to prove that f is a Hamiltonian quasi-Poisson map, we must still check that f∗ π1 = π2 , or, equivalently, that df π1 df ∗ = π2 . By Proposition 3.20, it suffices to prove that, for β ∈ T ∗ M2 , Y = df π1 df ∗ (β) ∈ T M2 satisfies (3.39) (Y, C2∗ (β)) ∈ L2 and dJ2 (Y ) = −(ρ2 σ ∨ )∗ β. Since f is an f-Dirac map, the first condition in (3.39) holds since (π1 df ∗ (β), df ∗ (C2∗ (β))) = (π1 df ∗ (β), C1∗ (df ∗ (β))) ∈ L1 ,

for L1 corresponds to π1 . The second condition holds since dJ2 (df π1 df ∗ (β)) = dJ1 (π1 df ∗ (β)) = −(ρ1 σ ∨ )∗ df ∗ (β) = −(ρ2 σ ∨ )∗ (β).

We now proceed to the proofs of Propositions 3.19 and 3.20. 3.5.2 Proofs Proof of Proposition 3.19. To simplify our formulas, we set T = ρM ρ ∨ dJ, and we denote by ·, · the pairing between vector spaces and their duals. First, we have to show that s(ξ ), r(ξ ) is antisymmetric in ξ, ξ ∈ A = T ∗ M ⊕g. We check this on elements of type (α, 0), (β, 0), and we leave the other cases to the reader. Since π is antisymmetric, we only have to show that T ∗ β, π (α) is antisymmetric in α and β. Using that dJ π = −(σ ∨ )∗ (ρM )∗ , which is the adjoint of the moment map condition (3.22), we see that ∗ ∗ (β), ρ ∨ (σ ∨ )∗ ρM (α), π(α, T ∗ β) = T ∗ β, π (α) = −ρM

(3.40)

which is antisymmetric by (3.29). We now turn to proving that s satisfies (3.5). For sections of A of type ξ = (0, u), ξ = (0, v), with u, v ∈ g, (3.5) follows from the next lemma. Lemma 3.25. Given a g-manifold M and an equivariant map J : M −→ G, then, for any u, v ∈ g, J ∗ σ ([u, v]) = LρM (u) (J ∗ σ (v)) − LρM (v) (J ∗ σ (u)) + dJ ∗ σ (v), ρM (u) − iρM (u)∧ρM (v) (J ∗ φ G ).

22


Proof. Using the equivariance of J , dJρM = ρ, we immediately see that this equation is the pullback by J of (3.5) for σ (for instance, the last term in the equation equals J ∗ iu∧v (φ G )).

Next we consider the case ξ = (0, u) and ξ = (α, 0), which is handled by the next result. Lemma 3.26. Given a g-manifold M, an equivariant map J : M −→ G, and a bivector π on M satisfying the moment map condition (3.22), then, for all v ∈ g and α ∈ T ∗ M, C ∗ LρM (v) (α) = LρM (v) (C ∗ (α)) − Lπ (α) (J ∗ σ (v)) + dJ ∗ σ (v), π (α) − iρM (v)∧π (α) (J ∗ φ G ). Although Lemma 3.26 is more difficult than Lemma 3.25, it is still simpler than the next case, treated in Lemma 3.27 below. Since a formula that holds under the same assumptions and is proved by the same method is proved in detail in Claim 3.37 below, we will omit its proof. Let us now consider ξ = (α, 0) and ξ = (β, 0). Comparing with Lemmas 3.25 and 3.26, the greater technical difficulty of this case comes from the fact that now the formulas involve both χG and φ G , the bracket [·, ·] induced by π on 1-forms, and require more than just the moment map condition. Lemma 3.27. Given a g-manifold M, an equivariant map J : M −→ G, and an invariant bivector π on M satisfying the moment map condition (3.22), then, for all α, β ∈ T ∗ M, 1 C ∗ ([α, β]) + J ∗ σ (i(ρM )∗ (α∧β) χG ) 2 = Lπ (α) C ∗ (β) − Lπ (β) C ∗ (α) − dC ∗ (β), π (α) − iπ (α)∧π (β) (J ∗ φ G ). Proof. Since C = 1 − 14 T , using the definition of s and of the bracket in (A), we see that we can rewrite the equation in the lemma as T ∗ ([α, β]) − Lπ (α) (T ∗ (β)) + Lπ (β) (T ∗ (α)) + dπ(α, T ∗ (β)) = 2J ∗ σ iρM∗ (α)ρM∗ (β) χG + 4iπ (α)∧π (β) J ∗ (φ G ).

(3.41)

Let us evaluate all the terms of (3.41) on an arbitrary vector field X ∈ X (M). To simplify the formulas, we set ∗ a = ρM (α),

∗ b = ρM (β),

V = J (X)

and we consider the Hom(g∗ , g)-valued function on G given by D = ρ ∨ (σ ∨ )∗ .

(3.42)


23

Claim 3.28. The following formula holds: dπ(α, T ∗ (β)), X = a, LV (Db) − b, LV (Da) − a, LV (D)b.

(3.43)

Proof. The left-hand side of (3.43) is LX π(α, T ∗ β). Hence, using (3.40), it equals ∗ ∗ ∗ ∗ (β), ρ ∨ (σ ∨ )∗ ρM (α) − ρM (β), LdJ (X) (ρ ∨ (σ ∨ )∗ )ρM (α). −LJ (X) ρM

(3.44)

With the notation of (3.42), and using D ∗ = −D (i.e. (3.29)) to rewrite the first term, we see that (3.44) equals DLV (b), a − b, LV (Da). To obtain (3.43), we write DLV (b) = LV (Db) − LV (D)(b).

From the definition of [α, β] (2.4), we have T ∗ ([α, β]) = T ∗ Lπ (α) (β) − T ∗ Lπ (β) (α) − T ∗ dπ(α, β).

(3.45)

Claim 3.29. The following formula holds: T ∗ dπ(α, β), X = π(LT (X) (α), β) + π(α, LT (X) (β)).

(3.46)

Proof. This follows from the invariance of π and the fact that the image of T sits inside that of ρM .

Using (3.45) and (3.46), we can split the left-hand side of (3.41) as a difference of two terms which are symmetric to each other. The next claim deals with such a term. Claim 3.30. The following formula holds: T ∗ Lπ (α) (β) − Lπ (α) (T ∗ (β)), X = π(LT (X) (α), β) + b, LV (Da) + b, dρ ∨ ((σ ∨ )∗ (a), V ).

(3.47)

Proof. The left-hand side of (3.47) equals −β, [π (α), T (X)] + T ([π (α), X]).

(3.48)

To rewrite [π (α), T (X)], we note that [π (α), ρM (v)] ˜ = −π LρM (v) ˜ ˜ (α) + ρM Lπ (α) (v),

(3.49)

for all v˜ ∈ C ∞ (M, g): Indeed, due to C ∞ (M)-linearity with respect to v, ˜ it suffices to check (3.49) for v˜ constant; in this case, the equation is just the invariance of π . We now use (3.49) for v˜ = ρ ∨ J (X) to get [π (α), T (X)] = −π LT (X) (α) + ρM Lπ (α) (ρ ∨ dJ (X)). We deduce that (3.48) equals

24

H. Bursztyn and M. Crainic ∗ ∗ β, π LT (X) (α) − ρM (β), Lπ (α) (ρ ∨ dJ (X)) + ρM (β), ρ ∨ J [π (α), X] ∗ (β), Lπ (α) (ρ ∨ J )(X). = π(LT (X) (α), β) − ρM

(3.50)

On the other hand, for all vector fields Y on M and g-valued 1-forms ν on G, we have iX LY (J ∗ ν) = LdJ (X) (ν(dJ (Y ))) + (dν)(dJ (Y ), dJ (X)). Using this identity for Y = π α and ν = ρ ∨ in (3.50), together with the dual of the moment map condition, dJ π = −((σ )∨ )∗ (ρM )∗ , we obtain (3.47) and prove the claim.

Combining the formulas of Claims 3.28, 3.29, and 3.30, we conclude that the left-hand side of (3.41) evaluated at a vector field X is b, dρ ∨ ((σ ∨ )∗ a, V ) − a, dρ ∨ ((σ ∨ )∗ b, V ) − a, LV (D)b.

(3.51)

On the other hand, the right-hand side of (3.41) applied to X equals ∗ ∗ 2(χG (ρM (α), ρM (β), σ ∗ dJ (X)) + 4φ G (dJ π (α), dJ π (β), dJ (X)))

= 2(χG (a, b, σ ∗ V ) + 4φ G ((σ ∨ )∗ a, (σ ∨ )∗ b, V )),

(3.52)

where we have used again that dJ π = −((σ )∨ )∗ (ρM )∗ . To conclude the proof of the lemma, it suffices to show that χG and φ G are related as follows. Claim 3.31. For all a, b ∈ g∗ and all vector fields V on G, one has 1 χG (a, b, σ ∗ V ) + φ G ((σ ∨ )∗ a, (σ ∨ )∗ b, V ) 2 1 = −a, dρ ∨ ((σ ∨ )∗ b, V ) + b, dρ ∨ ((σ ∨ )∗ a, V ) − a, LV (D)b . (3.53) 4 Proof. It suffices to prove (3.53) on elements of type a = u∨ , b = v ∨ , V = wr , where u, v, w ∈ g, and we recall that u∨ ∈ g∗ denotes the dual of u with respect to the quadratic form, and wr is the vector field on G obtained from w by right translations. We will also denote by Ad(u) ∈ C ∞ (G, g) the function g → Ad g (u), and we define Ad −1 (u) similarly. We will need the explicit formulas for σ ∗ and (σ ∨ )∗ : σ ∗ (wr ) =

1 (w + Ad −1 (w))∨ , 2

(σ ∨ )∗ (u∨ ) =

1 (ur + ul ). 2

Using these formulas, combined with the invariance of χG and φ G , the formula ul = Ad(ur ), and the explicit formulas for χG and φ G on elements of g, one can check that the left-hand side of (3.53) is


1 ([u, v], w + Ad −1 (w))g + ([u + Ad(u), v + Ad(v)], w)g . 8

25

(3.54)

Since ρ ∨ is the difference between the right and left Maurer–Cartan forms on G, we have (dρ ∨ )(ur , vr ) = −[u, v] − Ad −1 [u, v]. By the invariance of (·, ·)g with respect to Ad, we get that a, dρ ∨ ((σ ∨ )∗ b, V ) = −

1 (u, [v, w] + Ad −1 ([v, w]))g 2 + (u, [Ad(v), w] + [v, Ad −1 (w)])g

1 = − ([u + Ad(u), v + Ad(v)], w)g . 2

(3.55)

Since D = 12 (Ad − Ad −1 ), and Lwr (D)(v) = [w, Ad(v)] + Ad −1 ([w, v]), it follows that 1 a, LV (D)b = ([u, Ad(v)], w)g + ([Ad(u), v], w)g . 2 Hence the right-hand side of (3.53) equals 1 2([u + Ad(u), v + Ad(v)], w)g − ([u, Ad(v)], w)g − ([Ad(u), v], w)g , 8 which is easily seen to coincide with (3.54). This concludes the proof of the claim. Using Claim 3.31, we conclude that (3.51) and (3.52) coincide, and this proves Lemma 3.27.

From Lemmas 3.25, 3.26 and 3.27, it follows that s is a −J ∗ φ G -IM form for A. To conclude that L = Im(r, s) is a Dirac structure, we must still prove that L has rank n = dim(M). This follows from the next lemma (which also serves as inspiration for the proof of Proposition 3.20). Lemma 3.32. The sequence j

(r,s)

0 −→ T ∗ G −→ A −→ L −→ 0 is exact, where j (a) = (−J ∗ a, σ ∨ (a)), a ∈ T ∗ G. Proof. The fact that (r, s) ◦ j = 0 is equivalent to (3.22) and the second formula in (3.31). We define the maps U : A −→ T ∗ G, i : L −→ A,

1 ∗ U (α, v) = − (ρ ∨ )∗ ρM (α) + σ (v), 4 1 ∨ i(X, α) = α, ρ dJ (X) . 4

(3.56) (3.57)

26


We claim that U ◦ j = Id,

(r, s) ◦ i = Id,

and j ◦ U + i ◦ (r, s) = Id,

(3.58)

and these identities imply that the sequence is exact. For the first identity in (3.58), write 1 ∗ ∗ U (j (a)) = ρ ∨ ρM J a + σ σ ∨ a, 4 and then, using that dJρM = ρ and (3.26), we see that U ◦ j = Id. The second identity is immediate from the first and the last ones. To prove the last identity, we evaluate j (U (α, v)). The first component gives 1 ∨ ∗ ∗ 1 ∗ ∗ ∨ ∗ −J − (ρ ) ρM (α) + σ (v) = −J σ (v) + α − 1 − (ρM ρ J ) α 4 4 ∗ ∗ = −(J σ (v) + C (α)) + α. (3.59) The second component is

1 ∗ σ ∨ − (ρ ∨ )∗ ρM α + σ (v) . 4

(3.60)

∗ = −ρ ∨ (σ ∨ )∗ ρ ∗ = ρ ∨ dJ π , where we used (3.29) and the moment But σ ∨ (ρ ∨ )∗ ρM M map condition (3.22). Expressing σ ∨ σ using (3.25), we see that (3.60) is

1 v − ρ ∨ dJ (ρM (v) + π (α)). 4 Hence

1 ∨ j (U (α, v)) = (α, v) − s(α, v), ρ dJ r(α, v) , 4

i.e., j ◦ U + i ◦ (r, s) = Id. This concludes the proof of Proposition 3.19.

Proof of Proposition 3.20. Let J : (M, L) → (G, LG ) be a Dirac realization. Identifying LG with g G, we know that there is an induced action of g on M, denoted by ρM . Spelling out the definition, for v ∈ g, ρM (v) is the unique vector field satisfying the equations in (3.33). From the second condition in (3.33) and the fact that L is isotropic, we immediately deduce the following. Lemma 3.33. For all (X, α) ∈ L, ∗ ρM (α) + σ ∗ dJ (X) = 0.

Inspired by Lemma 3.32, we prove the following. Lemma 3.34. There is an exact sequence i

U

0 −→ L −→ T ∗ M ⊕ g −→ T ∗ G −→ 0, where U and i are given by (3.56) and (3.57), respectively.

(3.61)


27

Proof. First of all, U is surjective since, as in Lemma 3.32 (and keeping the same notation), U ◦ j = Id. Next, U ◦ i = 0 is an immediate consequence of (3.28) and (3.61). Finally, using the nondegeneracy condition (3.19) for a Dirac realization, it follows that i is injective. By a dimension argument, it follows that the sequence is exact.

We now concentrate on constructing the quasi-Poisson bivector field π . Following (ii) of Proposition 3.20, we have the following. Claim 3.35. π is well defined. Proof. We first show that (3.34) and (3.35) have a solution X, for any given α: the point is that the element 1 ∨ ∨ ∗ ∗ ∗ −C (α), ρ (σ ) ρM (α) 4 is in the kernel of U ; this is a simple computation using (3.26) and (3.29). Hence it must be in the image of i. More explicitly, we find that there exists an X such that ∗ (X, C ∗ (α)) ∈ L, ρ ∨ (dJ (X) + (σ ∨ )∗ ρM (α)) = 0.

(3.62)

On the other hand, applying Lemma 3.33 to (X, C ∗ (α)), and then using the first equation in (3.31) to replace CρM , we find that ∗ σ ∗ (dJ (X) + (σ ∨ )∗ ρM (α)) = 0.

(3.63)

Since Ker(σ ∗ ) ∩ Ker(ρ ∨ ) = 0, equations (3.62) and (3.63) imply (3.34). The uniqueness of X follows from the nondegeneracy condition (3.19).

Claim 3.36. π defines a bivector field π which satisfies the moment map condition (3.22). Proof. We have to show that α(π (β)) + β(π (α)) = 0 for all 1-forms α and β. Let X = π (α) and Y = π (β). Using (3.35) for (α, X) and (β, Y ), the fact that L is isotropic, and the definition of C, we find that 4(α(Y ) + β(X)) = α(ρM ρ ∨ dJ (Y )) + β(ρM ρ ∨ dJ (X)).

(3.64)

Let us show that the right-hand side of (3.64) is zero: using (3.34), (3.64) becomes α(ρM ρ ∨ (ρM σ ∨ )∗ (β)) + β(ρM ρ ∨ (ρM σ ∨ )∗ (α)), and this is zero due to (3.29). On the other hand, (3.34) shows that dJ π = −(ρM σ ∨ )∗ ; dualizing it (and using (π )∗ = −π , which holds by the first part of the lemma), we obtain the moment map condition.

28


Claim 3.37. The bivector field π is g-invariant. Proof. We have to show that LρM (v) (π (α)) = π (LρM (v) (α)) for v ∈ g, and 1-forms α. For this, it suffices to show that LρM (v) (π (α)) satisfies (3.34) and (3.35), i.e., dJ (LρM (v) (π (α))) = −(ρM σ ∨ )∗ LρM (v) (α), ∗

(LρM (v) (π (α)), C LρM (v) (α)) ∈ L.

(3.65) (3.66)

These conditions are related to Lemma 3.26. Let us first prove (3.66). Using (3.35), (3.33), and the fact that L is isotropic, we conclude that ([ρM (v), π (α)], LρM (v) (C ∗ α) − Lπ (α) (J ∗ σ (v)) + dJ ∗ σ (v), π (α) − iρM (v)∧π (α) (J ∗ φ G )) ∈ L. Using Lemma 3.26, we see that this expression is precisely (LρM (v) (π (α)), C ∗ LρM (v) (α)). Formula (3.65) is closely related to the one in Lemma 3.26: the proofs are similar and hold under the same hypothesis (which might be a bit surprising since (3.65) says that, although the invariance condition on π is not assumed, it must be satisfied modulo the kernel of J ). Since we have omitted the proof of Lemma 3.26, we will give the details for (3.65). We evaluate both sides of (3.65) on an arbitrary 1-form µ ∈ 1 (G). The left-hand side gives J ∗ µ, [ρM (v), π (α)] = d(J ∗ µ)(ρM (v), π (α)) + LρM (v) J ∗ µ, π (α) − Lπ (α) J ∗ µ, ρM (v) ∗ ∗ (α)) − LρM (v) µ, (σ ∨ )∗ ρM (α) = −(dµ)(ρ(v), (σ ∨ )∗ ρM + L(σ ∨ )∗ ρM∗ (α) µ, ρ(v). (3.67)

Evaluating µ on the right-hand side, we get −LρM (v) (α), ρM σ ∨ µ = −LρM (v) α, ρM σ ∨ µ + α, [ρM (v), ρM σ ∨ µ]. Now, using [ρM (v), ρM (v)] ˜ = ρM ([v, v]) ˜ + ρM LρM (v) (v) ˜ for v˜ = σ ∨ µ ∈ ∞ C (M, g), we get ∗ ∗ ∗ −LρM (v) ρM (α), σ ∨ µ + ρM (α), [v, σ ∨ µ] + ρM (α), LρM (v) (σ ∨ µ).

(3.68)

We have to show that this coincides with the r.h.s. of (3.67). Comparing the two ∗ α replaced by any formulas, we see that the resulting equation makes sense for ρM element in C ∞ (M, g∗ ). On the other hand, since the equation is C ∞ (M)-linear with respect to this element, we may assume that the element is a constant a ∈ g∗ (and the remaining appearances of ρM become ρ). The identity to be proved, relating the r.h.s. of (3.67) and (3.68), becomes −(dµ)(ρ(v), (σ ∨ )∗ a) − Lρ(v) µ, (σ ∨ )∗ a + L(σ ∨ )∗ a µ, ρ(v) = a, [v, σ ∨ µ],


or, equivalently,

−µ([ρ(v), (σ ∨ )∗ a]) = a, [v, σ ∨ µ].

29

(3.69)

We may assume that µ is the dual (with respect to the quadratic form) of the vector field wr for some w ∈ g, and that a is the dual of an element u ∈ g. Equation (3.69) becomes (after multiplying by 2): −(wr , [vr − vl , ur + ul ]) = (u, [v, w + Ad −1 (w)]), and this can be proved to hold from the invariance of the quadratic form and the identities [vl , ul ] = −[v, u]l (see (4.1) for the convention), [vr , ul ] = [vl , ur ].

Claim 3.38. The bivector field π is a quasi-Poisson tensor. Proof. We must show that π ([α, β]) = [π (α), π (β)] + 12 iα∧β (ρM (χG )). Using the definition of π ((ii) of Proposition 3.20) evaluated at [α, β], we have to show that 1 J [π (α), π (β)] + iα∧β (ρM (χG ) = −(ρM σ ∨ )∗ [α, β], (3.70) 2 1 ∗ (3.71) [π (α), π (β)] + iα∧β (ρM (χG )), C ([α, β]) ∈ L. 2 Similar to the discussion in the previous claim, these conditions are related to Lemma 3.27. The first equation holds under the same assumptions, and it is proved by the same method, so it will be left to the reader. (Similar to the discussion in the previous proof, the equation tells us that, although the quasi-Poisson condition is not assumed, it must be satisfied modulo the kernel of J .) We now prove (3.71). First, we use that (π (α), C ∗ (α)) ∈ L, (π (β), C ∗ (β)) ∈ L, the fact that L is isotropic, and then apply the formula in Lemma 3.27, to conclude that 1 [π (α), π (β)], C ∗ ([α, β]) − J ∗ σ iρM∗ (α∧β) (χG ) ∈ L. (3.72) 2 On the other hand, applying the action in (3.33) to v = iρM∗ (α∧β) (χG ) and observing that ρM (v) = iα∧β (ρM (χG )), we find that (iα∧β (ρM (χG )), J ∗ σ iρM∗ (α∧β) (χG )) ∈ L. Since L, at each point, is a vector space, (3.72) and (3.73) imply (3.71).

(3.73)

4 Moment maps in Dirac geometry: The global picture 4.1 Integrating Lie algebroids and infinitesimal actions Lie groupoids are the global counterparts of Lie algebroids. In order to fix our notation, we recall that a Lie groupoid over a manifold M consists of a manifold G together with

30


surjective submersions t, s : G → M, called target and source, a partially defined multiplication m : G (2) → G, where G (2) := {(g, h) ∈ G × G | s(g) = t(h)}, a unit section ε : M → G and an inversion G → G, all related by the appropriate axioms; see, e.g., [8]. To simplify our notation, we will often identify an element x ∈ M with its image ε(x) ∈ G. For a Lie groupoid G, the associated Lie algebroid A(G) consists of the vector bundle ker(ds)|M → M, (4.1) with anchor ρ = dt : ker(ds)|M → T M and bracket induced from the Lie bracket on X (G) via the identification of sections (ker(ds)|M ) with right-invariant vector fields on G tangent to the s-fibers. An integration of a Lie algebroid A is a Lie groupoid G together with an isomorphism A ∼ = A(G). Unlike Lie algebras, not every Lie algebroid admits an integration, see [14] for a description of the obstructions. On the other hand, if a Lie algebroid is integrable, then there exists a canonical source-simply-connected integration G(A); see [14]. If M is a point, then a Lie groupoid over M is a Lie group, and the associated Lie algebroid is its Lie algebra. Example 4.1 (transformation Lie groupoids). Let G be a Lie group acting from the left on a manifold M. The associated transformation Lie groupoid , denoted by GM, is a Lie groupoid over M with underlying manifold G × M, source map s(g, x) = x, target map t(g, x) = g · x, and multiplication (g, x) · (g , x ) = (gg , x ). In this case, A(G M) = g M, the transformation Lie algebroid associated with the infinitesimal action of g on M corresponding to the given G-action. (However, even if a g-action does not come from a global action of a Lie group, one can always find a Lie groupoid integrating the transformation Lie algebroid g M; see [16, 26].) Similar to infinitesimal actions, Lie groupoids act on maps into their identity sections: if G is a Lie groupoid over M, then a (left) action of G on a map J : N → M is a map mN : G ×M N → N , (g, y) → g · y, satisfying 1. J (g · y) = t(g), 2. (gg )y = g(g y), 3. J (y) · y = y. Here G ×M N := {(g, y) ∈ G × N | s(g) = J (y)}. For reasons that will be clear in the next two subsections, the map J : N → M is often referred to as the moment map of the action mN [25]. Example 4.2 (actions of transformation Lie groupoids). Analogous to Example 3.7, an action mN of a transformation Lie groupoid G = G M on a map J : N → M is equivalent to an ordinary action mN of the Lie group G on N for which J is G-equivariant. Indeed, mN and mN are related by mN ((g, J (y)), y) = mN (g, y),

where g ∈ G

and

y ∈ N.

(4.2)


31

The link between infinitesimal and global actions is based on the following notion: An infinitesimal action ρN of a Lie algebroid A is called complete if ρN (ξ ) ∈ X (N ) is a complete vector field whenever ξ ∈ (A) has compact support. As in the case of Lie algebras, a complete action of a Lie algebroid A can be integrated to an action of its canonical source-simply-connected integration G(A); see, e.g., [26]. 4.2 Poisson maps as moment maps for symplectic groupoid actions A 2-form ω on a Lie groupoid G is called multiplicative if the graph of the groupoid multiplication m : G (2) → G is an isotropic submanifold of (G, ω)×(G, ω)×(G, −ω). Equivalently, the multiplicativity condition for ω can be written as m∗ ω = pr ∗1 ω + pr ∗2 ω,

(4.3)

where pr i : G (2) → G, i = 1, 2, are the canonical projections. A symplectic groupoid [29] is a Lie groupoid together with a multiplicative symplectic form. Symplectic groupoids are the global counterparts of Poisson manifolds in the following sense: If π is a Poisson structure on a manifold P inducing an integrable Lie algebroid structure on A = T ∗ P (as in Section 2.2), then the associated sourcesimply-connected groupoid G(P ) := G(A) carries a natural multiplicative symplectic structure [9, 15, 23]; on the other hand, on any symplectic groupoid (G, ω) over a manifold P , condition (4.3) automatically implies that P has an induced Poisson structure uniquely determined by the condition that the target map t : G → P (respectively, source map s : G → P ) is a Poisson map (respectively, anti-Poisson map) [11]. An integration of a Poisson manifold (P , π) is a symplectic groupoid (G, ω) over P for which the induced Poisson structure coincides with π . Note that the symplectic form ω defines a vector bundle map ker(ds)|P −→ T ∗ P ,

ξ → iξ ω|T P ,

(4.4)

inducing an isomorphism of Lie algebroids A(G) ∼ = T ∗ P [11]. This immediately implies that dim(G) = 2 dim(P ). Example 4.3 (integrating Lie–Poisson structures). Let us consider g∗ , equipped with its Lie–Poisson structure. If G is a Lie group with Lie algebra g, then the transformation groupoid G = G g∗ , with respect to the coadjoint action, integrates T ∗ g∗ = g g∗ . The identification G × g∗ ∼ = T ∗ G by right translations induces a multiplicative symplectic form ω on G, in such a way that (G, ω) is a symplectic groupoid integrating g∗ . Remark 4.4. The construction of the symplectic groupoid in the previous example can be extended to the context of Poisson–Lie groups, see Remark 3.10: If (G, π ) is a simply connected Poisson–Lie group and G∗ is its dual, then, assuming that the dressing action is complete, the transformation groupoid G G∗ carries a symplectic structure making it into a symplectic groupoid integrating G∗ . (This symplectic

32


structure is basically the one associated with the semidirect product Poisson structure on G × G∗ induced from the action of G on itself by right multiplication.) For a more general construction when the actions are not complete, see [22]. Let us assume that P is an integrable Poisson manifold. We have seen that any Poisson map J : Q → P induces a Lie algebroid action of T ∗ P on Q. Analogous to the case of Lie algebras, when this action is complete, it can be “integrated’’ to an action of G(P ), the canonical source-simply-connected symplectic groupoid of P . We remark that the completeness of the T ∗ P action in the Lie algebroid sense coincides with the notion of J : Q → P being complete as a Poisson map, i.e., if f ∈ C ∞ (P ) has compact support (or if Xf is complete), then XJ ∗ (f ) is complete. The global action mN : G(P ) ×P Q → Q arising in this way is compatible with the Poisson structure on Q in the sense that graph(mN ) is a Lagrangian submanifold of (G(P ), π ) × (Q, πQ ) × (Q, −πQ ),3 where π is the Poisson structure associated with the symplectic form ω on G(P ). Since inclusions of symplectic leaves of Poisson manifolds are Poisson maps, an equivalent way to express this compatibility is that the restricted action mN : G(P ) ×P S → S to each symplectic leaf (S, ωS ) → (Q, πQ ) satisfies m∗N ωS = pr ∗G ω + pr ∗S ωS , (4.5) where pr G : G(P ) ×P S → G(P ) and pr S : G(P ) ×P S → S are the natural projections, see [25, 32]. On the other hand, if (Q, πQ ) is a Poisson manifold and mN is an action of a symplectic groupoid G on J : Q → P compatible with πQ in the sense just described, then J is automatically a Poisson map (this is just a leafwise version of [25, Thm. 3.8]). The next example is the global version of Example 3.8. Example 4.5 (global Hamiltonian actions). Consider g∗ with its Lie–Poisson structure, and let G be the simply connected Lie group with Lie algebra g. As in Example 3.8, the starting point is a Poisson map J : Q → g∗ . Note that J is complete as a Poisson map if and only if the associated infinitesimal g-action is by complete vector fields. In this case, the global action of the symplectic groupoid T ∗ G ∼ = G g∗ is equivalent, in the sense of Example 3.7, to the Hamiltonian G-action obtained by integrating the infinitesimal Hamiltonian g-action on Q. So, in the previous example, the “moment’’ J : Q → g∗ for the symplectic groupoid action of T ∗ G∗ is just a momentum map for a Hamiltonian G-action in the ordinary sense. Remark 4.6. Analogous to the previous example and following Remarks 3.10 and 4.4, a Poisson map J : Q → G∗ , where G∗ is the dual group to a complete simply connected Poisson Lie group, can be “integrated’’ to an action of the symplectic groupoid G G∗ , which is equivalent to a G-action on Q for which J is equivariant 3 A submanifold C of a Poisson manifold (P , π) is Lagrangian if, at each x ∈ P , the intersection of Tx C with π (Tx∗ P ), the tangent space to the symplectic leaf at x, is a Lagrangian subspace of π (Tx∗ P ).


33

(with respect to the dressing action on G∗ ). The “moment’’ J in this case coincides with Lu’s momentum map [21] for a Poisson action of a Poisson–Lie group on a Poisson manifold. 4.3 Dirac realizations as moment maps for presymplectic groupoid actions In order to describe the global actions “integrating’’ Dirac realizations, we should first identify the global objects integrating Dirac manifolds, generalizing symplectic groupoids. This was done in [6]: if φ is a closed 3-form on M, then a φ-twisted presymplectic groupoid over M is a Lie groupoid G over M equipped with a multiplicative 2-form ω such that 1. dω = s∗ φ − t∗ φ, 2. dim(G) = 2 dim(M), 3. ker(ωx ) ∩ ker(dx s) ∩ ker(dx t) = {0}, for all x ∈ M. (Twisted presymplectic groupoids are called quasi-symplectic groupoids in [33].) The multiplicativity of ω and condition 1 in this definition guarantee that the map σω : A → T ∗ M, ξ → iξ ω|T M

(4.6)

is a φ-IM form for A, while 2 and 3 are the extra conditions needed in Lemma 3.3 to insure that the image L of (ρ, σω ) is a φ-twisted Dirac structure. When (G, ω) is a symplectic groupoid, such L is precisely the Dirac structure associated with the induced Poisson structure on M. As proved in [6], L is uniquely determined by the condition that t is an f-Dirac map (respectively, s is an anti-f-Dirac map). Conversely, the canonical groupoid G(L) integrating the Lie algebroid associated with a φ-twisted Dirac structure (assuming it is integrable) is naturally a φ-twisted presymplectic groupoid [6, Sec. 5]. This correspondence generalizes the one between Poisson manifolds and symplectic groupoids [9, 15, 23] (see also [10] for the integration of twisted Poisson structures). We now have all the ingredients to generalize the “integration’’ procedure of Poisson maps to symplectic groupoid actions, explained in Section 4.2, to the context of Dirac geometry. Let LM be a φ-twisted Dirac structure on M associated with an integrable Lie algebroid. We call a Dirac realization J : N → M complete if the induced Lie algebroid action of LM on N is complete, in which case it integrates to an action mN : G(LM ) ×M N → N , where (G(LM ), ω) is the canonical twisted presymplectic groupoid associated with LM . In this situation, we will simply say that the action mN integrates the realization J . Theorem 4.7. Let (M, LM ) be a φ-twisted Dirac manifold and assume that LM is integrable. A complete Dirac realization J : N → M integrates to an action mN : G(LM ) ×M N → N satisfying m∗N LN = τpr∗G ω (pr ∗N LN ),

(4.7)

where pr G and pr N are the projections from G(LN ) ×M N onto G(LN ) and N , respectively, and τpr∗G ω denotes a gauge transformation.

34


Conversely, if mN is an action of G(LM ) on J : N → M satisfying (4.7), then J is f-Dirac; if J also satisfies (3.19), then it is a Dirac realization whose integration is mN . In order to prove the theorem, we need the following result. Lemma 4.8. Let (M, LM ) be a φ-twisted Dirac manifold and assume that LM is integrable. Let mN : G(LM ) ×M N → N be an action of G(LM ) on J : N → M, and assume that N is equipped with a J ∗ φ-twisted presymplectic form ωN . Then J is an f-Dirac map if and only if m∗N ωN = pr ∗N ωN + pr ∗G ω.

(4.8)

Proof. To simplify the notation, let G = G(LM ), and let us denote by A the corresponding Lie algebroid (which is just LM ). The source and target maps in G are denoted by s and t. Also, let ω1 = m∗N ωN − pr ∗N ωN and ω2 = pr ∗G ω. With these definitions, our goal is to show that J is f-Dirac if and only if ω1 = ω2 . The key observation is that if we regard G ×M N as a transformation Lie groupoid over N, with source pr N and target mN , a direct computation shows that both ω1 and ω2 are multiplicative. Hence, by [6, Thm. 2.5], ω1 = ω2 if and only if the corresponding bundle maps σωi : A ×M N → T ∗ N, ξy → σωi = (iξy ωi )|T N i = 1, 2, see (4.6), coincide. For ξy ∈ A ×M N (ξ ∈ Ax and x = J (y)) and Y ∈ T N (as usual, we identity T N with T ε(N ), where ε : N → G ×M N is the identity section), we have σω1 (ξy , Y ) = ωN (dmN (ξy ), Y ) and σω2 (ξy , Y ) = ω(ξ, dJ (Y )).

(4.9)

For the first identity in (4.9), we used that iξy pr ∗N ωN = 0 for ξy ∈ A ×M N , since pr N is the source map in G ×M N , and A ×M N is its Lie algebroid, which is tangent to the source fibres along the identity section. Since LM = {(dt(ξ ), iξ ω|T M ) | ξ ∈ A}, J : N → M being f-Dirac means that {(dt(ξ ), iξ ω|T M ) | ξ ∈ A} = {(dJ (Y ), α) | iY ωN = J ∗ α}.

(4.10)

But, for ξy ∈ A ×M N , we have dJ (dmN (ξy )) = dt(ξ ). It then follows from (4.10) that ω(ξ, dJ (Y )) = ωN (dmN (ξy ), Y ) for all Y ∈ T N, which implies that σω1 = σω2 , i.e., ω1 = ω2 . The converse follows from the same arguments, reversing the steps. We can now prove Theorem 4.7.


35

Proof. We keep writing G for G(LM ). Suppose that mN integrates a Dirac realization J : N → M. The bundles m∗N LN and pr ∗N LN , seen as subbundles of T (G ×M N ) ⊕ T ∗ (G ×M N ), have the same projection onto the first factor: at a point (g, y), they both coincide with Tg G × Ty O, where O is the leaf of LN through y. Note that, since pr N is a submersion, pr ∗N LN is a smooth subbundle, so it is an honest Dirac structure. By Corollary 3.13, since J is a Dirac realization of M, its restriction to any leaf of LN , (O, θ), is a presymplectic realization, and mN is tangent to the leaves. By Lemma 4.8, m∗N θ = pr ∗N θ + pr ∗G ω, which implies the compatibility (4.7). Conversely, (4.7) implies that J is tangent to the leaves of LN . Restricting mN to these leaves, (4.7) amounts to (4.8). So, by Lemma 4.8, J is an f-Dirac map when restricted to each leaf, which implies that J is f-Dirac by Corollary 3.6. The last statement follows from Corollary 3.13 and a direct check.

Remark 4.9. The presymplectic groupoid actions resulting from presymplectic realizations are exactly the “modules’’ considered in the Morita theory developed in [33] to compare various notions of moment maps. More general Dirac realizations give rise to more general “Hamiltonian spaces’’ which still fit with the constructions in [33]. We will discuss examples of the “integration’’ in Theorem 4.7 related to “quasi’’Hamiltonian actions in Section 4.5. 4.4 Reduction in Dirac geometry As in Poisson geometry, one can also carry out reduction in the context of Dirac manifolds. The general construction described in this section recovers reduction procedures in various settings, including [2, 3, 25, 33]. The setup is as follows. Let J : N → M be a Dirac realization of a φ-twisted Dirac manifold (M, LM ). Let x ∈ M be a regular value of J , and consider the submanifold ι : C = J −1 (x) → N . Following [25, 33], let lx = ker(ρ)x be the isotropy Lie algebra of LM at x. Since the anchor ρ is the projection pr 1 |LM , it follows that lx = (LM ∩ T ∗ M)x .

(4.11)

The induced Lie algebroid action of LM on J : N → M defines a vector bundle morphism LM ×M N → T N, and a simple computation shows that this morphism gives rise to an action of the Lie algebra lx on C. Our object of interest is the orbit space C/lx . Lemma 4.10. If the stabilizer algebras of the lx -action on C have constant dimension (on each component), then ι∗ LN is a (untwisted) Dirac structure on C. Proof. As mentioned in Section 3.2, the conclusion in the lemma holds as long as we show that ι∗ LN is a smooth subbundle of T C ⊕ T ∗ C. As a vector bundle, ι∗ LN is naturally identified with

36


LN ∩ (T C ⊕ T ∗ N ) , (LN ∩ T C ◦ )

(4.12)

see [12], and ι∗ LM will be smooth if we show that both bundles in (4.12) are smooth. For this, it suffices to show that each one has constant dimension. But since their quotient ι∗ LN has constant dimension, it suffices to show that either LN ∩(T C⊕T ∗ N ) or LN ∩ T C ◦ has constant dimension. We will prove that for LN ∩ T C ◦ . On the one hand, LN ∩ T C ◦ = {(0, β) ∈ LN | ι∗ β = 0} = {(0, dJ ∗ α) ∈ LN | α ∈ T ∗ M}. It follows from J being an f-Dirac map that if (0, dJ ∗ α) ∈ LN , then (0, α) ∈ LM . So, if ρN is the infinitesimal action of LM on J , we can write ker(ρN ) ∩ LM ∩ T ∗ M LN ∩ T C ◦ = {(0, dJ ∗ α) ∈ LN | α ∈ T ∗ M} ∼ . = ker(dJ ∗ ) But ker(ρN ) ∩ LM ∩ T ∗ M is the stabilizer of the lx -action on C, which is assumed to have constant dimension. Since x is a regular value, dJ has maximal rank on C, so ker(dJ ∗ ) also has constant dimension. As a result, the dimension of (4.12) is constant, and ι∗ LN is a smooth bundle. Finally, note that ι∗ LN is a (ι∗ J ∗ φ)-Dirac structure on C, but ι∗ J ∗ φ = 0. So ι∗ LN is an ordinary Dirac structure.

We now show that the quotient C/lx carries a natural Poisson structure. Theorem 4.11. Suppose that the orbit space C/lx is a smooth manifold so that projection C −→ C/lx is a submersion. Then there is a unique Poisson structure πred on C/lx for which the projection (C, ι∗ LN ) → (C/lx , πred ) is an f-Dirac map. Remark 4.12. The projection (C, ι∗ LN ) → (C/lx , πred ) is also a b-Dirac map, and this property characterizes πred uniquely as well. Proof. It follows from our assumptions that the lx -orbits on C have constant dimension, so the same holds for the stabilizer algebras. By Lemma 4.10, (C, ι∗ LN ) is a Dirac manifold. The admissible functions on (C, ι∗ LN ), i.e., the set of functions on C whose differential vanish on ker(ι∗ LN ) = ι∗ LN ∩ T C form a Poisson algebra (see [12, Sec. 2.5]) under the bracket {f, g} := LXf g, where Xf is a local vector field such that (Xf , df ) ∈ ι∗ LN . We will show that this Poisson algebra induces a Poisson structure on C/lx by showing that the kernel of ι∗ LN coincides with the lx -orbits, i.e., ker(ι∗ LN ) = ρN (lx ). On the one hand,

(4.13)


37

ι∗ LN ∩ T Q = {Y ∈ T Q | ∃β ∈ T ∗ N with (Y, β) ∈ LN , ι∗ β = 0} = {Y ∈ T Q | ∃α ∈ T ∗ M with (Y, dJ ∗ α) ∈ LN }. But since J is f-Dirac and dJ (Y ) = 0, we can write ι∗ LN ∩ T Q = {Y ∈ T Q | ∃α ∈ LM ∩ T ∗ M with (Y, dJ ∗ α) ∈ LN }. On the other hand, ρN (lx ) = {Y ∈ T N | ∃α ∈ LM ∩ T ∗ M with (Y, dJ ∗ α) ∈ LN , dJ (Y ) = 0} = {Y ∈ T Q | ∃α ∈ LM ∩ T ∗ M with (Y, dJ ∗ α) ∈ LN }. So (4.13) follows. The fact that the projection (C, ι∗ LN ) → (C/lx , πred ) is an f-Dirac map and the claim in Remark 4.12 follow from a direct computation; see, e.g., [7].

Of course, if the Dirac realization J : N → M is complete, one can state Theorem 4.11 in terms of the action of the isotropy group of G(LM ) at x ∈ M on C = J −1 (x). Versions of Theorem 4.11 can also be derived when this action is locally free and the quotient is an orbifold, as well as for more general “intertwiner spaces’’ in the sense of [33]. Remark 4.13 (other reductions). The following are important particular cases of the reduction in Theorem 4.11: •

•

•

If M is Poisson and J : N → M is a symplectic realization, we recover [25, Thm. 3.12]; in particular, when M = g∗ , this reduces to the Marsden–Weinstein classical theorem [24], and when M = G∗ , the dual of a Poisson–Lie group, we get Lu’s reduction [21]. If J : N → M is a Poisson map, we get the “Poisson version’’ of these results. If M is φ-twisted Dirac and J : N → M is a presymplectic realization, then we obtain Xu’s reduction [33, Thm. 3.17]; in particular, when M is a Lie group equipped with Cartan–Dirac structure, one recovers the quasi-Hamiltonian reduction of [3]. If J : N → G is a general Dirac realization of a Lie group with Cartan–Dirac structure, then we recover the reduction of quasi-Poisson manifolds of [2] via the identification established in Theorem 3.16; see Remark 4.16 below.

4.5 AMM-groupoids and Hamiltonian quasi-Poisson G-manifolds We now discuss global actions, in the sense of Theorem 4.7, associated with complete Dirac realizations of Cartan–Dirac structures. Let G be a Lie groups equipped with a Cartan–Dirac structure LG with respect to a bi-invariant nondegenerate quadratic form (·, ·)g . The first step is to identify G(LG ), the canonical presymplectic groupoid integrating LG .

38


As shown in [6, Sec. 7], G(LG ) is closely related to the AMM-groupoids of [5]: if G = G G is the transformation groupoid with respect to the conjugation action, then the 2-form [3] ω(g,x) =

1 (Ad x pg∗ λ, pg∗ λ)g + (pg∗ λ, px∗ (λ + λ))g , 2

where pg , px : G × G → G are the first and second projections, and λ and λ are the left and right Maurer–Cartan forms, makes G into a φ G -twisted presymplectic groupoid. If G is simply connected, then (G, ω) is isomorphic to G(LG ), the canonical source-simply-connected integration of LG . In general, G(LG ) is obtained from the G, where G is the universal cover of G [6, AMM groupoid by pulling back ω to G Thm. 7.6]. As a result, just as Lie–Poisson structures “integrate’’ to cotangent bundles of Lie groups, see Example 4.3, Cartan–Dirac structures “integrate’’ to the “double’’ (G × G, ω) in the sense of [3]. For simplicity, let G be simply connected. A complete Dirac realization J : M → G induces a presymplectic groupoid action of (G, ω), as in Theorem 4.7, which is equivalent to a G-action on M for which J is G-equivariant, see Example 4.2; this Gaction is just an integration of the infinitesimal g-action which makes M into a quasiPoisson g-manifold, as constructed in Proposition 3.20. So M becomes a Hamiltonian quasi-Poisson G-manifold for which J : M → G is the group-valued moment map [2]. This construction yields the following global version of Theorem 3.16. Theorem 4.14. There is a one-to-one correspondence between complete Dirac realizations of (G, LG ) and Hamiltonian quasi-Poisson G-manifolds. Corollary 4.15. There is a one-to-one correspondence between compact Dirac realizations of (G, LG ) and compact Hamiltonian quasi-Poisson G-manifolds. Of course, a global version of Proposition 3.24 also holds. Remark 4.16 (reduction). Given a Dirac realization of (G, LG ), J : M → G, the Dirac reduction of Theorem 4.11 produces Poisson spaces J −1 (g)/Gg , where Gg is the centralizer of g ∈ G. Using Remark 4.13 and [2, Prop. 10.6], one can check that these are the same Poisson spaces obtained by quasi-Poisson reduction [2, Thm.6.1] if we regard M as a Hamiltonian quasi-Poisson G-manifold instead. Acknowledgments We would like to thank many people for helpful discussions concerning this work, including A. Alekseev, Y. Kosmann-Schwarzbach, E. Meinrenken, D. Roytenberg, A. Weinstein, P. Xu, and the referees. Our collaboration was facilitated by invitations to the conferences “PQR2003,’’ in Brussels, and “AlanFest’’ and “Symplectic Geometry and Moment Maps,’’ held at the Erwin Schrödinger Institute, where most of the results in this paper were announced; we thank the organizers of these meetings, in particular A. Alekseev, S. Gutt, J. Koiller, J. Marsden, and T. Ratiu. For financial support, H. B. thanks DAAD (German Academic Exchange Service) and M. C. thanks KNAW (Dutch Royal Academy of Arts and Sciences). H. B. thanks Freiburg University for its hospitality while part of this work was being done.


39

References [1] A.Alekseev and Y. Kosmann-Schwarzbach, Manin pairs and moment maps, J. Differential Geom., 56 (2000), 133–165. [2] A. Alekseev, Y. Kosmann-Schwarzbach, and E. Meinrenken, Quasi-Poisson manifolds, Canadian J. Math., 54 (2002), 3–29. [3] A. Alekseev, A. Malkin, and E. Meinrenken, Lie group valued moment maps, J. Differential Geom. 48 (1998), 445–495. [4] M. Bangoura and Y. Kosmann-Schwarzbach, The double of a Jacobian quasi-bialgebra, Lett. Math. Phys., 28 (1993), 13–29. [5] K. Behrend, P. Xu, and B. Zhang, Equivariant gerbes over compact simple Lie groups, C. R. Acad. Sci. Paris, 336 (2003), 251–256. [6] H. Bursztyn, M. Crainic, A. Weinstein, and C. Zhu, Integration of twisted Dirac brackets, Duke Math. J., 123-3 (2004), 549–607. [7] H. Bursztyn and O. Radko, O, Gauge equivalence of Dirac structures and symplectic groupoids, Ann. Inst. Fourier (Grenoble), 53 (2003), 309–337. [8] A. Cannas da Silva and A. Weinstein, Geometric Models for Noncommutative Algebras, American Mathematical Society, Providence, RI, 1999. [9] A. Cattaneo and G. Felder, Poisson sigma models and symplectic groupoids, in Quantization of Singular Symplectic Quotients, Progress in Mathematics, Vol. 198, Birkhäuser, Basel, 2001, 61–93. [10] A. Cattaneo and P. Xu, Integration of twisted Poisson structures, J. Geom. Phys., 49-2 (2004), 187–196. [11] A. Coste, P. Dazord, and A. Weinstein, Groupoïdes symplectiques, in Publications du Département de Mathématiques. Nouvelle Série A, Vol. 2, i–ii, Université Claude-Bernard, Lyon, 1987, 1–62. [12] T. Courant, Dirac manifolds, Trans. Amer. Math. Soc., 319 (1990), 631–661. [13] T. Courant and A. Weinstein, Beyond Poisson Structures, Séminaire sud-rhodanien de géométrie VIII, Travaux en Cours, Vol. 27, Hermann, Paris, 1988, 39–49. [14] M. Crainic and R. Fernandes, Integrability of Lie brackets, Ann. Math., 157 (2003), 575–620. [15] M. Crainic and R. Fernandes, Integrability of Poisson Brackets, Math.DG/ 0210152. [16] P. Dazord, Groupoïde d’holonomie et géométrie globale, C. R. Acad. Sci. Paris, 324 (1997), 77–80. [17] K. Guruprasad, J. Huebschmann, L. Jeffrey, andA. Weinstein, Groups systems, groupoids, and moduli spaces of parabolic bundles, Duke Math. J., 89 (1997), 377–412. [18] P. Higgins and K. Mackenzie, Algebraic constructions in the category of Lie algebroids, J. Algebra, 129 (1990), 194–230. [19] C. Klimˇcik and T. Ströbl, WZW-Poisson manifolds, J. Geom. Physics, 4 (2002), 341–344. [20] J.-H. Lu, Multiplicative and Affine Poisson Structures on Lie Groups, Ph.D. thesis, University of California at Berkeley, Berkeley, 1990. [21] J.-H. Lu, Momentum mappings and reduction of Poisson actions, in Symplectic Geometry, Groupoids, and Integrable Systems (Berkeley, CA, 1989), Springer-Verlag, New York, 1991, 291–311. [22] J.-H. Lu and A. Weinstein, Groupoïdes symplectiques double des groupes de Lie-Poisson, C. R. Acad. Sci. Paris, 309 (1989), 951–954. [23] K. Mackenzie and P. Xu, Integration of Lie bialgebroids, Topology, 39 (2000), 445–467. [24] J. Marsden and A. Weinstein, Reduction of symplectic manifolds with symmetry, Rep. Mathematical Phys., 5 (1974), 121–130.

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[25] K. Mikami and A. Weinstein, Moments and reduction for symplectic groupoid actions, Publ. RIMS Kyoto Univ., 24 (1988), 121–140. [26] I. Moerdijk and J. Mrˇcun., On integrability of infinitesimal actions, Amer. J. Math., 124 (2002), 567–593. [27] J.-S. Park, Topological open p-branes, in Symplectic geometry and Mirror symmetry (Seoul 2000), World Scientific Publishing, River Edge, NJ, 2001, 311–384. [28] P. Ševera and A. Weinstein, Poisson geometry with a 3-form background, Progr. Theoret. Phys. Suppl., 144 (2001), 145–154. [29] A. Weinstein, Symplectic groupoids and Poisson manifolds, Bull. Amer. Math. Soc. (N.S.), 16 (1987), 101–104. [30] A. Weinstein, Poisson geometry. Symplectic geometry, Differential Geom. Appl., 9 (1998), 213–238. [31] A. Weinstein, The geometry of momentum, in Proceedings of the Conference on “Geometry in the 20th Century: 1930–2000,’’ to appear; Math.SG/0208108. [32] P. Xu,Morita equivalent symplectic groupoids, in Symplectic Geometry, Groupoids, and Integrable Systems (Berkeley, CA, 1989), Springer-Verlag, New York, 1991, 291–311. [33] P. Xu, Morita Equivalence and Momentum Maps, preprint; Math.SG/0307319.

Construction of Ricci-type connections by reduction and induction∗ Michel Cahen1 , Simone Gutt1,2 , and Lorenz Schwachhöfer3 1 Université Libre de Bruxelles

Campus Plaine, CP 218 BE-1050 Brussels Belgium [email protected] 2 Université de Metz Ile du Saulcy F-57045 Metz Cedex 01 France [email protected] 3 Mathematisches Institut Universität Dortmund Vogelppothsweg 87 D-44221 Dortmund Germany [email protected] It is a pleasure to dedicate this paper to Alan Weinstein on the occasion of his 60th birthday. Abstract. Given the Euclidean space R2n+2 endowed with a constant symplectic structure and the standard flat connection, and given a polynomial of degree 2 on that space, Baguis and Cahen [1] have defined a reduction procedure which yields a symplectic manifold endowed with a Ricci-type connection. We observe that any symplectic manifold (M, ω) of dimension 2n (n ≥ 2) endowed with a symplectic connection of Ricci type is locally given by a local version of such a reduction. We also consider the reverse of this reduction procedure, an induction procedure: we construct globally on a symplectic manifold endowed with a connection of Ricci type (M, ω, ∇) a circle or a real line bundle which embeds in a flat symplectic manifold (P , µ, ∇ 1 ) as the zero set of a function whose third covariant derivative vanishes in such a way that (M, ω, ∇) is obtained by reduction from (P , µ, ∇ 1 ). We further develop the particular case of symmetric symplectic manifolds with Ricci-type connections.

∗ This research was partially supported by an Action de Recherche Concertée de la Commu-

nauté française de Belgique.

42

M. Cahen, S. Gutt, and L. Schwachhöfer

1 Introduction A symplectic connection ∇ on a symplectic manifold (M, ω) of dimension 2n is a linear connection which is torsion free and for which ω is parallel. The space of symplectic connections on (M, ω) is infinite dimensional. Selecting some particular class of connections by curvature conditions has, a priori, two interests. The “moduli space’’ of such particular connections may be finite dimensional and, on some compact symplectic manifolds which do admit a connection of the chosen class, this connection may be “rigid.’’ In this paper, we describe completely the local behavior of symplectic connections of Ricci type (see definition below) and give some global description of simply connected symplectic manifolds admitting a connection of Ricci type. We denote by R the curvature of ∇ and by R the symplectic curvature tensor R(X, Y, Z, T ) := ω(R(X, Y )Z, T ). For any point x ∈ M, we have the symmetry properties (i) R x (X, Y, Z, T ) = −R x (Y, X, Z, T ) (ii) R x (X, Y, Z, T ) = R x (X, Y, T , Z) (iii) + R x (X, Y, Z, T ) = 0. X,Y,Z

From (i) and (ii), R x ∈ 2 Tx∗ M ⊗ 2 Tx∗ M, where k V is the symmetrized ktensor product of the vector space V . We denote by r the Ricci tensor of the connection ∇ (i.e., rx (X, Y ) = tr [Z → Rx (X, Z)Y ], where X, Y, Z are in Tx M); this tensor r is symmetric. We denote by ρ the corresponding endomorphism of the tangent bundle ω(X, ρY ) := r(X, Y ) so that ρx belongs to the symplectic algebra sp(Tx M, ωx ) and tr ρ = 0. The space Rx of symplectic curvature tensors at x is Rx = ker a ⊂ 2 Tx∗ M ⊗ 2 Tx∗ M, where a is the skew-symmetrization map a : p Tx∗ M ⊗ q Tx∗ M → p+1 Tx∗ M ⊗ q−1 Tx∗ M a(u1 ∧ · · · ∧ up ⊗ v1 . . . vq ) :=

q

u1 ∧ · · · ∧ up ∧ vi ⊗ v1 . . . vî . . . vq .

i=1

The group Sp(Tx M, ωx ) acts on Rx . Under this action the space Rx , in dimension 2n ≥ 4, decomposes into two irreducible subspaces [6], Rx = Ex ⊕ Wx , and the decomposition of the curvature tensor R x into its Ex component (denoted Ex ) and its Wx component (denoted Wx ), R x = Ex + Wx , is given by

Construction of Ricci-type connections by reduction and induction

Ex (X, Y, Z, T ) = −

43

1 2ωx (X, Y )rx (Z, T ) + ωx (X, Z)rx (Y, T ) 2(n + 1)

+ ωx (X, T )rx (Y, Z) − ωx (Y, Z)rx (X, T ) − ωx (Y, T )rx (X, Z) . A connection ∇ is said to be of Ricci type if, at each point x, Wx = 0. (Let us mention that such connections were called reducible by Vaisman in [6].) In dimension 2 (n = 1), the space W vanishes identically. We shall assume in what follows that the manifold has dimension m = 2n > 2. Let us first recall two interesting features of such connections. •

When a symplectic connection is of Ricci type, it satisfies the equations + (∇X r)(Y, Z) = 0.

X,Y,Z

•

Those are the Euler–Lagrange equations of any natural variational principle whose Lagrangian is a second degree invariant polynomial in the curvature (r 2 or R 2 ). Connections which are solutions of those equations are called preferred. They are completely described in dimension 2. The condition to be of Ricci type is the condition on a symplectic connection ∇ to have an integrable almost complex structure J ∇ on the twistor space over M which is the bundle of all compatible almost complex structures on M [2].

In this paper, we show that any symplectic manifold (M, ω) of dimension 2n (n ≥ 2) admitting a symplectic connection of Ricci type has a local model given by a reduction procedure (as introduced by Baguis and Cahen in [1]) from the Euclidean space R2n+2 endowed with a constant symplectic structure and the standard flat connection. We also consider the reverse of this reduction procedure, an induction procedure: we construct globally on a simply connected symplectic manifold endowed with a connection of Ricci type (M, ω, ∇) a circle or a real line bundle N which embeds in a flat symplectic manifold (P , µ, ∇ 1 ) as the zero set of a function whose third covariant derivative vanishes in such a way that (M, ω, ∇) is obtained by reduction from (P , µ, ∇ 1 ). We finally describe completely the symmetric symplectic manifolds whose canonical connection is of Ricci type. Those were already studied in [4] in collaboration with John Rawnsley.

2 Some properties of the curvature of a Ricci-type connection Let (M, ω) be a smooth symplectic manifold of dim 2n (n ≥ 2) and let ∇ be a smooth Ricci-type symplectic connection. The following results follow directly from the definition (and Bianchi’s second identity). Lemma 2.1 ([3]). The curvature endomorphism reads

44


R(X, Y ) = −

1 [−2ω(X, Y )ρ −ρY ⊗X +ρX ⊗Y −X ⊗ρY +Y ⊗ρX], (1) 2(n + 1)

where X denotes the 1-form i(X)ω ( for X a vector field on M) and where, as before, ρ is the endomorphism associated with the Ricci tensor [r(U, V ) = ω(U, ρV )]. Furthermore, (i) there exists a vector field u such that ∇X ρ = −

1 [X ⊗ u + u ⊗ X]; 2n + 1

(2)

(ii) there exists a function f such that ∇X u = −

2n + 1 2 ρ X + f X; 2(n + 1)

(3)

(iii) there exists a real number K such that trρ 2 +

4(n + 1) f = K. 2n + 1

(4)

3 Construction by reduction of manifolds with Ricci-type connections Let A be a nonzero element in the symplectic Lie algebra sp(R2n+2 , ), where is the standard symplectic structure on R2n+2 . Let A be the closed hypersurface A ⊂ R2n+2 with equation (5)

(x, Ax) = 1; in order for A to be nonempty we replace, if necessary, A by −A. Let ∇˙ be the standard flat symplectic affine connection on R2n+2 . If X, Y are vector fields tangent to A , define A (∇X Y )(x) = (∇˙ X Y )(x) − (AX, Y )x;

(6)

this is a torsion free linear connection on A . The vector field Ax is an affine vector field for this connection; it is clearly complete and we denote by φt the 1-parametric group of diffeomorphisms of A generated by this vector field; clearly this flow is given by the restriction to A of the action of exp tA on R2n+2 . Since the vector field Ax is nowhere 0 on A , for any x0 ∈ A , there exists • • • •

a neighborhood Ux0 (⊂ A ), a ball D ⊂ R2n of radius r0 , centered at the origin, a real interval I = (−, ), and a diffeomorphism χ : D × I → Ux0 such that χ (0, 0) = x0 and χ (y, t) = φt (χ (y, 0)).

(7)


We shall denote π : Ux0 → D,

45

π = p1 ⊗ χ −1 .

If we view A as a constraint manifold in R2n+2 , D is a local version of the Marsden– Weinstein reduction of A around the point x0 . If x ∈ A , Tx A =Ax⊥ , where v1 , . . . , vp denotes the subspace spanned by v1 , . . . , vp and ⊥ denotes the orthogonal relative to ; let Hx (⊂ Tx A ) =x, Ax⊥ ; then Tx R2n+2 = (Hx ⊕ RAx) ⊕ Rx and π∗x defines an isomorphism between Hx and the tangent space Ty D for y = π(x). A vector belonging to Hx will be called horizontal. A symplectic form on D, ω, is defined by ¯ Y¯ ), ωy (X, Y ) = x (X,

y = π(x),

(8)

where X¯ (respectively, Y¯ ) denotes the horizontal lift of X (respectively, Y ). A symplectic connection ∇ on D is defined by A ¯ ¯ ¯ ∇X Y (x) = ∇X ¯ Y (x) + (X, Y )Ax.

(9)

Proposition 3.1 ([1]). The manifold (D, ω) is a symplectic manifold and ∇ is a symplectic connection of Ricci type. Furthermore, a direct computation shows that the corresponding ρ, u and f are given by ¯ ρX(x) = −2(n + 1)Ax X, u(x) ¯ = ∗

−2(n + 1)(2n + 1)A2x x, 2

(π f )(x) = 2(n + 1)(2n + 1) (A x, Ax),

(10) (11) (12)

where Akx is the map induced by Ak with values in Hx : Akx (X) = Ak X + (Ak X, x)Ax − (Ak X, Ax)x.

4 Local models for symplectic connections of Ricci type The properties of a symplectic connection of Ricci type, as stated in Lemma 2.1, imply in particular that • • • •

the curvature tensor is determined by ρ; its covariant derivative is determined by u; its second covariant derivative is determined by ρ and f , hence by ρ and K with K a constant; the third covariant derivative of the curvature is determined by u, ρ, K, and similarly for all orders. Hence we have the following.

46


Corollary 4.1. Let (M, ω) be a smooth symplectic manifold of dimension 2n (n ≥ 2) and let ∇ be a smooth Ricci-type connection. Let p0 ∈ M; then the curvature Rp0 and its covariant derivatives (∇ k R)p0 (for all k) are determined by (ρx0 , ux0 , K). Corollary 4.2. Let (M, ω, ∇) (respectively, (M , ω , ∇ )) be two real analytic symplectic manifolds of the same dimension 2n (n ≥ 2), each endowed with a real analytic symplectic connection of Ricci type. Assume that there exists a linear map b : Tx0 M → Tx0 M such that (i) b∗ ωx = 0

ωx0 ; (ii) bux0 = u x ; (iii) b ◦ ρx0 ◦ b−1 = ρx . Assume further that K = K . 0 0 Then the manifolds are locally affinely symplectically isomorphic, i.e., there exists a normal neighborhood of x0 (respectively, x0 ), Ux0 (respectively, Ux ), and a sym0

plectic affine diffeomorphism ϕ : (Ux0 , ω, ∇) → (Ux , ω , ∇ ) such that ϕ(x0 ) = x0 0 and ϕ∗x0 = b.

This follows from classical results, see for instance Theorem 7.2 and Corollary 7.3 in Kobayashi–Nomizu Vol. 1 [5]. Consider now (M, ω, ∇) a real analytic symplectic manifold of dimension 2n (n ≥ 2) endowed with an analytic Ricci-type symplectic connection; denote as before by u, ρ, f and K the associated quantities (see Lemma 2.1). Let p0 be a point in M and choose ξ0 a symplectic frame of Tp0 M, i.e., a linear symplectic isomorphism ξ0 : (R2n , ) → (Tp0 , ωp0 ), where is the standard symplectic form on R2n . Denote by u(ξ ˜ 0 ) the element of R2n corresponding to u(p0 ), i.e., u(ξ ˜ 0 ) = (ξ0 )−1 u(p0 ) and by ρ(ξ ˜ 0 ) the element of sp(R2n , ) corresponding to ρ(p0 ), i.e., ρ(ξ ˜ ) = (ξ0 )−1 ρ(p0 ) ξ0 . Define an element A of sp((R2n+2 , ) as ⎛ ⎞ −u(ξ ˜ 0) f (p0 ) ⎜ 0 2(n + 1)(2n + 1) 2(n + 1)(2n + 1) ⎟ ⎟ ⎜ ⎟ ⎜ 0 0 A = ⎜1 ⎟, ⎟ ⎜ ⎠ ⎝ −ρ(ξ ˜ 0) −u(ξ ˜ 0) 0 2(n + 1)(2n + 1) 2(n + 1) where u(ξ ˜ 0 ) = i(u(ξ ˜ 0 )) and where we have chosen a basis {e0 , e0 , e1 , . . . , e2n } of the symplectic vector space R 2n+2 relative to which the symplectic form has matrix ⎛ ⎞ 0 1 0 0 In ⎝ ⎠

= .

= −1 0 0 , −In 0 0 0 Consider the local reduction procedure described in Section 3 from the element A defined above around the point x0 = e0 ∈ A = {x ∈ R2n+2 | (x, Ax) = 1}.


47

From what we saw in Section 3 this yields a symplectic manifold with a Ricci-type connection (M , ω , ∇ ). Denote by π the map π : Ue0 → M , where Ue0 is the neighborhood of e0 in A ⊂ R2n+2 considered in Section 3 and consider y0 = π (e0 ). Then He0 = e0 , Ae0 = e0 ⊥ =e1 , . . . , e2n is isomorphic under π∗ to Ty0 M . Introduce the injection j : R2n → R2n+2 with j (x1 , . . . , x2n ) = (0, 0, x1 , . . . , x2n ) so that j (R2n ) = He0 and denote by b : Tp0 M → Ty0 M the map given by b = π∗ e ◦ j ◦ ξ0−1 . 0

This map b is a linear symplectic isomorphism since ωy 0 (bX, bY ) = (j ξ0−1 X, j ξ0−1 Y ) = (ξ0−1 X, ξ0−1 Y ) = ωp0 (X, Y ). Furthermore, u (y0 ) = π∗ e (u¯ (x0 )) 0

= π∗ e (−2(n + 1)(2n + 1)(A2 e0 − (A2 e0 , Ae0 )e0 )) 0

˜ 0 )) = π∗ e (ξ0 )−1 u(p0 ) = bu(p0 ) = π∗ e (j u(ξ 0

0

ρ (y0 )bX = π∗ e ρ (y0 )X(e0 ) = π∗ e (−2(n + 1)Ae0 (j ξ0−1 (X))) 0

=

0

˜ 0 )ξ0−1 (X)) π∗ e (j ρ(ξ 0

so that ρ (y0 )b = bρ(p0 ) (f )(y0 ) = 2(n + 1)(2n + 1) (A2 e0 , Ae0 ) = f (p0 ). Hence we have the following. Theorem 4.3. Any real analytic symplectic manifold with a Ricci-type connection is locally symplectically affinely isomorphic to the symplectic manifold with a Riccitype connection obtained by a local reduction procedure around e0 = (1, 0, . . . , 0) from a constraint surface A defined by a second order polynomial in the standard ˙ flat symplectic manifold (R2n+2 , , ∇).

5 Construction of a contact manifold which is a global circle or line bundle over M Consider (M, ω, ∇) a smooth symplectic manifold of dimension 2n > 2 with a π smooth Ricci-type connection and let B(M) → M be the Sp(R2n , )-principal bundle of symplectic frames over M. (An element in the fiber over a point p ∈ M is a symplectic isomorphism ξ : (R2n , ) → (Tp M, ωp )). As before, we consider u˜ : B(M) → R2n the Sp(R2n , ) equivariant function given by u(ξ ˜ ) = ξ −1 u(x) where x = π(ξ )

48


and ρ˜ : B(M) → sp(R2n , ) the Sp(R2n , ) equivariant function given by ρ(ξ ˜ ) = ξ −1 ρ(x)ξ and we define the Sp(R2n , ) equivariant map A˜ : B(M) → sp(R2n+2 , ) ⎛ ⎞ −u(ξ ˜ ) (π ∗ f )(ξ ) ⎜ 0 2(n + 1)(2n + 1) 2(n + 1)(2n + 1) ⎟ ⎟ ⎜ ⎟ ˜ )=⎜ 0 0 A(ξ ⎟, ⎜1 ⎟ ⎜ ⎠ ⎝ −ρ(ξ ˜ ) −u(ξ ˜ ) 0 2(n + 1)(2n + 1) 2(n + 1)

(13)

where V = i(V ) for V in R2n . We inject the symplectic group Sp(R2n , ) into Sp(R2n+2 , ) as the set of matrices I2 0 ˜ , A ∈ Sp(R2n , ). j (A) = 0 A Lemma 5.1. Define the 1-form α on B(M), with values in sp(R2n+2 , ) by ⎛ ⎞ ) −ρ(X)(ξ −ωx (u, X) ⎟ ⎜ 0 ⎜ 2(n + 1)(2n + 1) 2(n + 1) ⎟ ⎜ hor ˜ ) ⎟ ⎟, 0 0 −X(ξ αξ (X ) = ⎜ ⎟ ⎜ ⎟ ⎜ ⎠ ⎝ −ρ(X)(ξ ) ˜ 0 X(ξ ) 2(n + 1)

(14)

hor

where X ∈ Tx M with x = π(ξ ) and X is the horizontal lift of X in Tξ B(M), and by α(C ∗ ) = j˜∗ (C) (15) for all C ∈ sp(R2n , ), where C ∗ denotes the fundamental vertical vector field on d B(M) associated with C (Cξ∗ = dt ξ. exp tC|0 ). This form has the following properties: (i) Rh∗ α = Ad(j˜(h−1 ))α ∀h ∈ Sp(R2n , ); ˜ (ii) d A˜ = −[α, A]; ˜ ∗ ω. (iii) dα + [α, α] = −2Aπ p

When one has a G-principal bundle P → M, an embedding of the group G in a larger group G , j : G → G , and a 1-form α with values in the Lie algebra of G , such that α(C ∗ ) = j∗ (C) for all C in the Lie algebra of G and Rh∗ α = Ad(j (h−1 )) α for p

all h in G, one can build the G -principal bundle P = P ×G G → M and the unique connection 1-form on P , α satisfying i ∗ α = α, where i : P → P ; ξ → [(ξ, 1)]. In our situation we build the Sp(R2n+2 , )-principal bundle B (M) = B(M) ×Sp(R2n , ) Sp(R2n+2 , )


49

whose elements are equivalence classes of pairs (ξ, g), ξ ∈ B(M), g ∈ Sp(R2n+2 , ), with (ξ, g) equivalent to (ξ h, j˜(h−1 )g) ∀h ∈ Sp(R2n , ). The projection π : B(M) → M maps [(ξ, g)] to π(ξ ). The connection 1-form α is characterized by the fact that α[ξ,1] ([X

hor

, 0]) = αξ (X

hor

)

and the equations above give the following. Lemma 5.2. The curvature 2-form of the connection 1-form α is equal to −2A˜ π ∗ ω, where A˜ is the unique Sp(R2n+2 , )-equivariant extension of A˜ to B (M). This curvature 2-form is invariant by parallel transport (d α curv(α ) = 0). Thus the holonomy algebra of α is of dimension 1. Corollary 5.3. Assume M is simply connected. The holonomy bundle of α is a circle π

or a real line bundle over M, N → M. This bundle has a natural contact structure ν given by the restriction to N ⊂ B(M) of the 1-form −α (viewed as real valued since it is valued in a one-dimensional algebra). One has dν = 2π ∗ ω. It is enlightening to point out the link between the holonomy bundle N over M and the constraint surface A when one sees M as obtained (locally) by reduction. The link is only local since A is in general not a principal bundle over M; in fact in most cases the quotient of A by the action of the group exp tA is at best an orbifold. Let A be a nonzero element of sp(R2n+2 , ) and let A = {y ∈ R2n+2 |

(y, Ay) = 1}; we assume as before that it is not empty. Assume that (M, ω, ∇) is obtained by reduction from A (as before, we restrict ourselves to some open set in A ). Let y0 be a point in A , let x0 = π(y0 ) ∈ M and choose a symplectic frame ξ0 at x0 . Let γ (t) be a curve in M such that γ (0) = x0 . Let ξ(t) be the symplectic frame at γ (t) obtained by parallel transport along γ from ξ0 and let y(t) be the horizontal curve in A lifting γ (t) from y0 (i.e., π(y(t) = γ (t) and (y(t), y(t)) ˙ = 0). Define the element C(t) of Sp(R2n+2 , ) as the matrix whose columns are C(t) = (y(t) Ay(t) ξ(t)), where ξ(t) consists of the 2n vectors which are the horizontal lifts at the point y(t) of the vectors of the frame ξ(t) (the image under the map ξ(t) of the usual basis of R2n ). Then d hor C(t)|s = C(s).αξ(s) (γ˙ (s) ), dt hor

where α is the 1-form on B(M) defined in (14) and where X is the horizontal lift hor of X in B(M); hence γ˙ (s) = ξ˙ (s). Let B (M) be the Sp(R2n+2 , )-principal bundle over M considered above and let [(ξ0 , 0 )] (where 0 is an element in Sp(R2n+2 , )) be a point of B (M) above x0 . The horizontal lift of γ (t) to B (M) starting from [(ξ0 , 0 )] lives in the holonomy subbundle containing this point; it reads

50


[(ξ(t), D(t))], where ξ(t) has been defined above and where D(t) obeys the differential equation d D(t)|s = −αξ(s) (ξ˙ (s)).D(s) dt and has initial value 0 . Define the map above γ which sends y(t) to [(ξ(t), D(t))], where D(t) = C −1 (t)C(0)0 ; this map sends elements of A to elements in the holonomy bundle through [(ξ0 , 0 )]. The map from the holonomy bundle through [(ξ0 , 0 )] to R2n+2 given by [(ξ, D)] → C0 0 D −1 e0 , where C0 is a fixed element in Sp(R2n+2 , ) has value in the hypersurface A , ˜ 0 )C −1 . where A = C0 A(ξ 0

6 Embedding of the contact manifold in a flat symplectic manifold Let (M, ω) be a smooth symplectic manifold of dim 2n (n ≥ 2) and let ∇ be a smooth symplectic connection of Ricci type. Let (N, α) be a smooth (2n + 1)-dimensional contact manifold (i.e., α is a smooth 1-form such that α ∧(dα)n = 0 everywhere). Let X be the corresponding Reeb vector field (i.e., i(X)dα = 0 and α(X) = 1). Assume there exists a smooth submersion π : N → M such that dα = 2π ∗ ω. Then at each point x ∈ N, Ker(π∗x ) = RX and LX α = 0. Remark that such a contact manifold always exists if M is simply connected as we saw in the previous section. If U is a vector field on M we can define its “horizontal lift’’ U on N by (i) π∗ U = U , (ii) α(U ) = 0. Let us denote by ν the 2-form ν = dα = 2π ∗ ω on N . Define a connection ∇ N on N by ∇ N U V = ∇U V − ν(U , V )X 1 ∇N XU = ∇N U X = − ρU 2(n + 1) 1 ∇N XX = − u, 2(n + 1)(2n + 1) where ρ is the Ricci endomorphism of (M, ∇) and where u is the vector field on M appearing in ∇ρ; see Lemma 2.1. Then ∇ N is a torsion free connection on N and the Reeb vector field X is an affine vector field for this connection.


51

The curvature of this connection has the following form: 1 [ν(ρV , W )U − ν(ρU , W )V ] 2(n + 1) 1 R N (U , V )X = [ν(u, V )U − ν(u, U )V ] 2(n + 1)(2n + 1) 1 1 R N (U , X)V = ν(u, V )U + ν(U , ρV )X 2(n + 1)(2n + 1) 2(n + 1) 1 R N (U , X)X = [−π ∗ f U + ν(U , u)X], 2(n + 1)(2n + 1)

R N (U , V )W =

where f is the function appearing in Lemma 2.1. Consider now the embedding of the contact manifold N into the symplectic manifold (P , µ) of dimension 2n + 2, where P = N × R, and, if we denote by s the variable along R and let θ = e2s p1∗ α (p1 : P → N ), we set µ = dθ = 2e2s ds ∧ α + e2s dα and let i : N → P , x → (x, 0). Obviously, i ∗ µ = ν. We now define a connection ∇ 1 on P as follows. If Z is a vector field along N , we denote by the same letter the vector field on P such that (i) Zi(x) = i∗x Z, (ii) [Z, ∂s ] = 0. The formulas for ∇ 1 are ∇Z1 Z = ∇ N Z Z + γ (Z, Z )∂s , where γ (Z, Z ) = γ (Z , Z) 1 π ∗f γ (X, X) = 2(n + 1)(2n + 1) 1 γ (X, U ) = − ν(u, U ) 2(n + 1)(2n + 1) 1 γ (U , V ) = ν(U , ρV ), 2(n + 1) and ∇Z1 ∂s = ∇∂1s Z = Z ∇∂1s ∂s = ∂s .

52


Theorem 6.1. The connection ∇ 1 on (P , µ) is symplectic and has zero curvature. Proposition 6.2. Let ψ(s) be a smooth function on P . Then ψ has vanishing third covariant differential if and only if ∂s2 ψ − 2∂s ψ = 0.

(16)

In particular the function e2s has this property. The procedure described above is called the induction. Let (P , µ, ∇ 1 ) be as above and let = N be the constrained submanifold defined by e2s = 1. Let Y be the vector field transversal to such that i(Y )µ = α, thus Y = ∂s . Let H be the 1-parametric group generated by X. Then /H can be identified with M and (M, ω) is the classical Marsden–Weinstein reduction of (P , µ) for the constraint . The connection ∇ on M is obtained from the flat connection ∇ 1 on (P , µ) by reduction. Hence we have the following. Corollary 6.3. Any smooth simply connected symplectic manifold with a Ricci-type connection (M, ω, ∇) can be obtained by reduction from an hypersurface in a flat symplectic manifold (P , µ, ∇ 1 ) defined by the 1-level set of a function ψ on P whose third covariant derivative vanishes. Corollary 6.4. Any smooth simply connected symplectic manifold with a Ricci-type connection (M, ω, ∇) is automatically analytic. Proof. Since (P , µ, ∇ 1 ) is locally symmetric, P , µ and ∇ 1 are real analytic and the explicit construction given preserves analyticity.

7 Symmetric symplectic spaces with Ricci-type connections Lemma 7.1. The reduction construction described in Section 3 yields a locally symmetric symplectic space (i.e., such that the curvature tensor is parallel) if and only if the element 0 = A ∈ sp(R2n+2 , ) satisfies A2 = λI for a constant λ ∈ R. Proof. Indeed the connection ∇ has parallel curvature tensor if and only if ∇ρ = 0 hence iff u = 0. From the formulas above, this is true iff A2x (x) = A2 x − (A2 x, Ax)x = 0 for any x ∈ A . When u = 0, f is a constant (cf. Lemma 2.1) and it follows from Lemma 3.1 that (A2 x, Ax) is a constant λ. Since A contains a basis of R2n+2 , this yields A2 = λI .


53

Proposition 7.2. If 0 = A ∈ sp(R2n+2 , ) satisfies A2 = λI for a constant λ ∈ R, the quotient of A by the action of exp tA is a manifold and the natural projection map A → M is a submersion which endows A with a structure of circle or real line bundle over M. Proof. Consider 0 = A ∈ sp(R2n+2 , ) so that A2 = λI . Case 1: λ > 0, say λ = k 2 with k > 0. Then there exists a basis of R2n+2 in which kIn+1 0 0 In A= ,

= 0 −kIn+1 −In 0 so that A = {(u, v) u, v ∈ Rn+1 | −2ku · v = 1}. The flow of the vector field Ax is given by φt = etA . The map π : A → T S n = {(u , v ) u , v ∈ Rn+1 |u · u = 1, u · v = 0} defined by u u , u(v + π(u, v) = ) u 2ku2 induces a diffeomorphism between M = A /φt and T S n . M is a noncompact simply connected manifold and A is a R-bundle over T S n . Case 2: λ < 0, say λ = −k 2 with k > 0. One splits V C (V = R2n+2 ) into the eigenspaces relative to A, V C = Vik ⊕ V−ik and observe that those subspaces are Lagrangian. Choosing a basis {z1 , . . . , zn+1 } for Vik ωkl := (zk , zl ); then , consider i iω is a Hermitian matrix. A change of basis (zj = zi Uj ) yields ω =t U ωU so we can find a basis for Vik so that 0 Ip ω = −2iIp,n+1−p = −2i . 0 −In+1−p In the basis of R2n+2 given by ej = 12 (zj + zj ), fj = 2i1 (zj − zj ), we have 0 −kI 0 Ip,n+1−p A= ,

= kI 0 −Ip,n+1−p 0 so that A = {(u, v) u, v ∈ Rn+1 | k i≤p ((ui )2 +(v i )2 )−k i>p ((ui )2 +(v i )2 ) = ∼

1}. We assume p ≥ 1 or replace A by −A so that A = S 2p−1 × R2n−2p+2 is nonempty. The flow φt is given by the action of cos ktI − sin ktI exp tA = . sin ktI cos ktI Then M = A /φt = (S 2p−1 × R2n−2p+2 )/U (1), so this reduced manifold is • • •

M = R2n if p = 1; M is a complex line bundle of rank q := n + 1 − p over the complex projective space Pp−1 (C) = S 2p−1 /U (1) if 1 < p ≤ n; M = Pn (C) if p = n + 1.

In all those cases, M is simply connected and A is a circle bundle over M; the only compact case is M = Pn (C).

54


Case 3: λ = 0, so A2 = 0 with A = 0. Let us denote by p the rank of A. One splits V = R2n+2 into V = V0 ⊕ V1 ⊕ V2 , where V1 = Im A (dim V1 = p), V0 ⊕V1 = Ker A (so dim V0 = 2n+2−2p and V0 is symplectic, since V0 ⊕V1 = V1⊥ ) and V2 is a Lagrangian subspace of V0⊥ supplementary to V1 . Choose a basis of V2 and a corresponding basis (dual for ) in V1 and a symplectic basis of V0 so that in those basis ⎛ ⎞ ⎛ ⎞ 00 0

1 0 0 A = ⎝ 0 0 A ⎠ ,

= ⎝ 0 0 Ip ⎠ 00 0 0 −Ip 0 the basis and A is symmetric. Changing the basis of V2 and correspondingly of V1 , one can bring A to the form A = Ir,p−r so that (x, Ax) = i≤r (w i )2 − r 1 and A consists of two copies of R2n+1 if r = 1. The action of φt on (u, v, w) is given by φt (u, v, w) = (u, v + tA w, w) so the reduced manifold is • •

two copies of R2n (if r = 1); or M = S r−1 × R2n+1−r if r > 1.

In all cases, M is a noncompact manifold and A is a line bundle over M.

Proposition 7.3. If 0 = A ∈ sp(R2n+2 , ) satisfies A2 = λI for a constant λ ∈ R, the quotient manifold is a symmetric space and the connection obtained by reduction is the canonical symmetric connection. Proof. Any linear symplectic transformation B of R2n+2 which commutes with A obviously induces a symplectic affine transformation β(B) of the reduced space M = A /φt . If π denotes the canonical projection π : A → M, then β(B) ◦ π = π ◦ B. In particular the symmetry at the point x = π(y), y ∈ A is induced by By u = −u + 2 (u, Ay)y − 2 (u, y)Ay.

The list of all symmetric spaces whose canonical connection is of Ricci type and the fact that the only compact simply connected one is Pn (C) already appears in [4]. What we describe here is a construction of all those manifolds by global reduction from the flat Euclidean space. We shall now describe the transvection group of M (i.e., the group G of affine transformations of M generated by the composition of two symmetries). Let us denote by G the group G = {B ∈ Sp(R 2n+2 , ) | BA = AB}. The transvection group of M is clearly included in β(G ); in fact it is the smallest subgroup of β(G ) stable under conjugation by a symmetry and which acts transitively on M. Let x0 = π(y0 ) be a point in M and let sx0 = β(By0 ) be the symmetry at this point. Consider the automorphism of G given by conjugation by By0 and denote by σ the


55

induced automorphism of the Lie algebra g of G . Let p = {C ∈ g | σ (C) = −C} and k = {C ∈ g | σ (C) = C}. The dimension of p is equal to 2n. Indeed, in a basis {e0 , e0 , e1 , . . . , e2n } of 2n+2 R in which e0 = y0 and e0 = Ae0 and ⎛ ⎞ 0 1 0

= ⎝ −1 0 0 ⎠ , 0 0 one has

⎛ ⎞ ⎞ 0λ 0 10 0 A = ⎝1 0 0 ⎠, By0 = ⎝ 0 1 0 ⎠ , 0 0 A 0 0 −I2n ⎧⎛ ⎞ ⎨ b λc A Z g = ⎝ c −b −Z ⎠ , b, c ∈ R; Z ∈ R2n ; B ∈ sp(R2n , ) ⎩ Z A Z B ⎫ ⎬ such that BA = A B , ⎭ ⎛

and ⎫ ⎧⎛ ⎞ ⎬ ⎨ 0 0 A Z p = ⎝ 0 0 −Z ⎠ , Z ∈ R2n . ⎭ ⎩ Z A Z 0 Hence the Lie algebra of the transvection group is equal to β∗ (p + [p , p ]). In all cases the kernel of β is given by exp tA, and the transvection group is described as follows: Case 1: λ > 0, say λ = k 2 with k > 0. In the basis of R2n+2 in which 0 0 In kIn+1 ,

= A= , 0 −kIn+1 −In 0 we have G =

B 0 0 (t B)−1

, B ∈ Gl(n + 1, R) ,

and β of such an element is the identity iff B = λI with λ > 0. The transvection group G is isomorphic to Sl(n + 1, R) and T S n = Sl(n + 1, R)/ Gl(n, R). Case 2: λ < 0, say λ = −k 2 with k > 0. In the basis of R2n+2 in which 0 Ip,n+1−p 0 −kI , A= ,

= −Ip,n+1−p 0 kI 0

56


we have G =

B1 B 2 −B2 B1

, B1 + iB2 ∈ U (p, n + 1 − p) ,

and β of such an element is the identity iff B1 + iB2 = exp −ikt. The transvection group G is isomorphic to SU (p, n + 1 − p) and M = SU (p, n + 1 − p)/U (p − 1, n + 1 − p). Case 3: λ = 0, rank A = k = p + q. In the basis of R2n+2 in which ⎞ ⎛ 00 0 A = ⎝ 0 0 Ipq ⎠ 00 0 and ⎞

1 0 0

= ⎝ 0 0 −I ⎠ , 0 I 0 ⎛

we have

⎧⎛ ⎞ D 0 C ⎨ g = ⎝ −t C 1 −t B F ⎠ , D ∈ sp(R2n+2−2k , ω1 ), B ∈ so(p, q, R), ⎩ 0 0 B ⎫ ⎬ F ∈ gl(k, R), t F = F, C ∈ Mat(2n + 2 − 2k, k, R) . ⎭

Then p is given by the elements of g for which D = 0, C = CJ , F = −J F J , B = −J BJ , where 1 0 J = , 0 −Ik−1 so C = (u 0 . . . 0) for u ∈ R2n+2−2k ,

F = for v ∈ Rk−1 , and

B=

0 tv v 0

0 t w w 0

for w ∈ Rk−1 and w = Ip−1,q w. Hence p ⊕ [p , p ] is the set of all elements in g for which D = 0. The transvection group G has algebra g isomorphic to {(B, F, C)}/(0, RIpq , 0), where B is any element in so(p, q, R), F is any symmetric real k × k matrix, and C is any real (2n + 2 − 2k) × k matrix and the bracket is defined by


57

[(B, F, C), (B , F , C )] = ([B, B ], −t C 1 C +t C 1 C −t BF +t B F, CB − C B), so when p+q > 2, the Levi factor is so(p, q, R) and the radical is a two-step nilpotent algebra. If p = 0 and q = 1 the transvection group is R2n and the symmetric space is the standard symplectic vector space. If p = q = 1 or if p = 0 and q = 2, the transvection group is solvable but not nilpotent. The two solvable examples are interesting for building exact quantization.

References [1] P. Baguis and M. Cahen, A construction of symplectic connections through reduction, Lett. Math. Phys., 57 (2001), 149–160. [2] F. Burstall and J. Rawnsley, private communication; see also N. R. O’Brian and J. H. Rawnsley, Twistor spaces, Ann. Global Anal. Geom., 3 (1985), 29–58 and I. Vaisman, Variations on the theme of twistor spaces, Balkan J. Geom. Appl., 3 (1998), 135–156. [3] M. Cahen, S. Gutt, J. Horowitz, and J. Rawnsley, Homogeneous symplectic manifolds with Ricci-type curvature, J. Geom. Phys., 38 (2001), 140–151. [4] M. Cahen, S. Gutt, and J. Rawnsley, Symmetric symplectic spaces with Ricci-type curvature, in G. Dito and D. Sternheimer, eds., Conférence Moshé Flato 1999: Quantization, Deformations, and Symmetries, Vol. II, 1999, Mathematical Physics Studies, Vol. 22, Kluwer Academic Publishers, Dordrecht, The Netherlands, 2000, 81–91. [5] S. Kobayashi and K. Nomizu, Foundations of Differential Geometry, Vols. I and II, Wiley, New York, London, 1963. [6] I. Vaisman, Symplectic curvature tensors, Monats. Math., 100 (1985), 299–327; see also M. De Visher, Mémoire de Licence, Bruxelles, 1999.

A mathematical model for geomagnetic reversals J. J. Duistermaat Department of Mathematics Utrecht University Postbus 80 010 3508 TA Utrecht The Netherlands [email protected]

1 Introduction The earth’s magnetic field has reversed its polarity many times in history, where the polarity of the magnetic field remained the same for very long time intervals, between about one hundred thousand years and many million years, whereas the reversals took place in a relatively short time interval of the order of magnitude of a thousand years. The lengths of time intervals between the subsequent reversals form an irregular sequence with a large variation, which make the reversals look like a (Poisson) stochastic process; see [7]. The direction of the earth’s magnetic field has been recorded in the basalt rocks of the ocean floors and in sedimentary rocks. In the first case the alignment of the magnetic particles is frozen in the rock when the upwelling fluid-hot basalt at the mid-ocean ridges solidifies upon cooling and then is pushed aside by the subsequent upwelling. This leads to a fantastic zebra-like stripe pattern in the alignments of the magnetic material in the ocean floor, the discovery of which actually was one of the most convincing arguments for the concept of sea-floor spreading. Fixing alignment during sedimentation is another recording mechanism. Compared to the basaltic rocks, the historical record of the earth’s magnetic field in sedimentary rocks reveals more details about the shorter time scales, but become harder to interpret in the very old rocks because of the frequent deformations of the sedimentary material. Some years ago Peter Hoyng from SRON (an institute in Utrecht which puts astronomical instruments into satellites) came to me with a question about some partial differential equations, which turned out to be related to a mathematical model which Schmitt, Ossendrijver, and he had formulated for the reversals of the earth’s magnetic field in [4] and [5]. In their model, the earth’s magnetic field is supposed to be a solution of a stochastically perturbed dynamical system in which the unperturbed deterministic system has two competing stable equilibria. The domains of attraction are separated by the stable manifold of a saddle point at the origin, where the magnetic field is equal to zero. A typical feature of their model is that the stochastic perturbation is proportional to the magnetic field, and therefore its coefficients vanish at the origin.

60

J. J. Duistermaat

The vanishing of the stochastic term at the origin corresponds to the appearance of the factor B in the term αB in equation (1) in loc. cit., where the factor α contains the stochastic fluctuations. These fluctuations come from the superposition of a turbulent flow superimposed upon the main flow in the liquid outer core. Such turbulent perturbations have no accurate descriptions in terms of simple deterministic models, whereas simple stochastics models lead to reasonable agreement with observations of time averages of turbulent perturbations. In [5] the predictions of the model have been compared in detail with the data on the geomagnetic dipole moment, including the statistics of the reversals. Good, although not complete agreement was obtained and the conclusion in [5] is that the model is consistent with the data. Several groups have made three-dimensional magnetohydrodynamic simulations which looks very much earth-like, leading to a largely dipolar exterior field, about 0.5 G at the surface, and sudden reversals. However, the parameter regime of these simulations is still many orders of magnitude removed from reality. For example, the Ekman number (ratio of typical magnitude of viscous to Coriolis forces) is about 10−15 , but the simulations can only get down to 10−6 . The agreement therefore could be just accidental. Apart from this, we believe that there is merit in “simple’’ analytical models which might give insight into what goes on both in the simulations and in the earth. It should also be observed that in other astrophysical objects the behavior of the magnetic field can be very different. For instance, the magnetic field of the sun has a strong deterministic component which is periodic with a period of about 22 years instead of being stationary. Accordingly, the physical models of the sun are quite different from those of the earth. See, for instance, [9]. Let u(x) denote the expectation value of the first time of exit from one of the domains of attraction, for the stochastic process which starts at the point x ∈ . The function u(x) satisfies an elliptic inhomogeneous linear partial differential equation in the domain , with the Dirichlet boundary condition that u(x) = 0 when x ∈ ∂ . The problem is singularly perturbed because the assumption of the smallness of the stochastic perturbation of the deterministic system leads to a small positive coefficient in front of the second-order derivatives. Another complication is that the vanishing of the stochastic term at the origin implies that the differential operator is no longer elliptic at the origin, a point on the boundary of . Actually, if we replace the deterministic vector field by its linearization at the origin, then the stochastic process is invariant under homotheties, and the mean exit time would be constant on every ray in starting from the origin. This leads to discontinuous behavior at the origin, which we conjecture is inherited by the function u(x) in our nonlinear model. Other quantities, like the invariant probability measure (if it exists) satisfy similar singularly perturbed partial differential equations, which also degenerate at the origin. From my knowledge of partial differential equations, I could not answer Hoyng’s question about the asymptotic behavior of the solutions as the stochastic perturbation tends to zero. Instead, prompted by suggestions of the stochastic experts in our department, I tried to apply the theory of Freidlin and Wentzell [10, 2] concerning small stochastic perturbations of dynamical systems. It turned out that this could not be done directly, because their theory is about compact domains, whereas ours is not

A mathematical model for geomagnetic reversals

61

and, more importantly, our problem degenerates at the origin. Still, the arguments of the theory appear to carry through, although the full proof of this is not yet finished and will be the subject of a more extensive paper. In this paper I will confine myself to the description of the results which would follow from the properly extended theory of Freidlin and Wentzell. If the stochastic terms are of small order , then the probabilities turn out to be of 2 order e−c/ , in which c is some positive real number. Because ratios of such exponential expressions are again such exponential expressions, the asymptotics for the probabilities depend very sensitively on the value of the coefficient c. Such behavior is called large deviations.

2 The stochastic process The model consists of a stochastic differential equation dx(t) = dt · b(x(t)) +

k

dBj ◦ Xj (x(t)),

j =1

where the process x(t) is a curve in the configuration space M, which is assumed to be a smooth manifold. The b(x) and Xj (x), 1 ≤ j ≤ k, are vector fields on M, whereas dBj denote independent Brownian motions on the reals. The vector field b describes the deterministic dynamical system, whereas dBj ◦ Xj (x) is a Brownian motion proportional to the vector field Xj (x). The symbol ◦ indicates that we use the Stratonovich integral, in which the symmetric midpoint rule at subsequent time steps is used in the approximating Riemann sums. It leads to a coordinate invariant calculus on the manifold M; see [1, pp. 74, 75, 111–115], [6, pp. 100, 101, 233–235], or [8, pp. 24, 35–37], which is convenient when we make substitutions of variables. The expectation value u(x, t) of f (x(t)), under the condition that x(0) = x, satisfies the partial differential equation ∂u/∂t = Au,

u(x, 0) = f (x),

in which the second-order linear partial differential operator 1 2 Xj 2 k

A=b+

j =1

is called the infinitesimal generator of the process. Here the vector fields b and Xj are viewed as first-order linear partial differential operators. The probability distribution µ, giving a chance to arrive in a given subset at time t if one starts at the point x, satisfies the adjoint equation ∂µ/∂t = A∗ µ, where µ at t = 0 is equal to the Dirac measure at x. Here A∗ denotes the adjoint of the operator A acting on distributions.

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Because both the deterministic system and the stochastic perturbation have variable coefficients, one needs a priori estimates which ensure that the solutions of the stochastic differential equation exist with probability one for all time. Similarly, one needs a priori estimates for the existence of an invariant probability measure µ, i.e., a measure which satisfies the equation A∗ µ = 0, where the uniqueness of such a measure follows if the infinitesimal generator A is elliptic. The required a priori estimates can be obtained with the use of Lyapunov-like functions W which satisfy inequalities like AW ≤ −1 in the complement of a compact subset of M; see [3].

3 Large deviations If Xj (x) ∼ σj (x) for small , then the principal symbol of A is equal to 2 a(x)(ξ, ξ )/2, in which the inner product a(x) on covectors is defined by a(x)(ξ, η) =

k

σj (x), ξ · σj (x), η,

ξ, η ∈ (Tx M)∗ .

j =1

That is, the partial differential equations are singularly perturbed , which implies, among other things, that they are numerically unstable. The inner product a(x) induces an inner product g(x) = a(x)−1 on the tangent space at x, which defines a Riemannian structure on the manifold M. The theory of Freidlin and Wentzell [10], [2] states the following. For every smooth curve γ : [0, T ] → M, there exists a real number S(γ ) such that for every δ > 0 and η > 0, there exists an 0 > 0 with the following property. If p denotes the probability that the process x(t) which starts at γ (0) has the property that for every t ∈ [0, T ] the distance from x(t) to γ (t) does not exceed δ, then e−S(γ )+η)/ ≤ p ≤ e−(S(γ )−η)/ 2

2

whenever 0 < || ≤ 0 . The required smoothness is that γ should have a square integrable derivative, and the estimates are uniform when T remains bounded, γ remains in a compact subset of M and S(γ ) remains bounded. Here S(γ ) denotes the “action integral’’ 1 T S(γ ) = g(γ (t))(v(t), v(t))dt, 2 0 where we have written v(t) = γ (t) − b(γ (t)), and η > 0 is arbitrarily small. In other words, the coefficient in the exponent of the small deviations estimate is equal to one half of the integral of the square of the length of the difference between the actual velocity vector and the velocity vector of the deterministic system. Here the length of the tangent vector v at x, with respect to the Riemannian structure g, is equal to g(x)(v, v)1/2 . Of course, one could also include the factor 1/ 2 in the definition of the functional S, which would amount to replacing the Riemannian structure g by −2 g, or


63

replacing the expression a(x)(ξ, ξ )/2 by the principal symbol 2 a(x)(ξ, ξ )/2 of the infinitesimal generator A of the stochastic process. However natural this may be, we follow the custom of using a functional S which does not depend on , and write the factor 1/ 2 in the exponents of the asymptotic estimates of the probabilities. For quite general systems, Freidlin and Wentzell derived similar exponential estimates for the following: • • •

the probability that the process which starts at x leaves a given domain near a given point, the expectation value of the first time of exit from the domain, and the invariant probability distribution in the position space.

It is a great challenge for analysts to derive such estimates from the singularly perturbed partial differential equations which are satisfied by these quantities. Here “directly’’ would mean “without probabilistic arguments.’’ The results of Freidlin and Wentzell are described in terms of the two-point function V (x, y) = inf {S(γ ) | γ (0) = x, γ (T ) = y}, in which T is arbitrary. It can be proved that this function is Lipschitz continuous in all the variables. Let D be a relatively compact open subset of the domain of attraction of a stable equilibrium s of the deterministic system. Let E be the set of points of the boundary where V (s, z), z ∈ ∂D, is minimal. Then with overwhelming probability the process, which starts at any given point x ∈ D, will leave D near E. Moreover, again with overwhelming probability, the process, after leaving a small neighborhood of s for the last time, stays close to a minimizing curve from s to a point y ∈ E. As we will discuss in the next Section 4, such a curve is equal to the projection to the position space of a solution of the Hamiltonian system on the unstable manifold of (s, 0). Finally, the mean exit time from D is (asymptotically for 2 2 → 0) equal to eV (s,y)/ , modulo factors eη/ with arbitrarily small |η|. Note that because V (s, y) > 0, this means that the mean exit time is exponentially large when 2 is small.

4 A Hamiltonian system If the minimum is attained at a curve γ , then γ satisfies the Euler–Lagrange equations [L]i :=

d ∂L ∂L − = 0 in which x = γ (t), v = γ (t), dt ∂vi ∂xi

for the Lagrange function L(x, v) =

1 g(x)(v − b(x), v − b(x)). 2

Moreover, γ (t) and b(γ (t)) have the same g-length, meaning that

(4.1)

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g(x)(v, v)1/2 = g(x)(b(x), b(x))1/2

when x = γ (t), v = γ (t).

(4.2)

Via the Legendre transform, these minimizing curves correspond to the solutions (x(t), ξ(t)) of the Hamiltonian system defined by the function 1 H (x, ξ ) = b(x), ξ + a(x)(ξ, ξ ), 2 where, moreover, H (x(t), ξ(t)) ≡ 0.

(4.3)

Proof. The Legendre transform assigns to an arbitrary function L(x, v) of the position x and the velocity v the function H (x, ξ ) = v, ξ − L(x, v)

(4.4)

of the position x and the momentum vector ξ , in which v is expressed as a function v = v(ξ ) of ξ by means of the equations ∂L(x, v)/∂vi = ξi ,

1 ≤ i ≤ n.

(4.5)

The point is that the Euler–Lagrange equations [L] = 0 for the function L, which express that γ (t) is a stationary curve for the integral T S= L(γ (t), γ (t))dt, 0

are equivalent to the condition that (γ (t), ξ(t)) is a solution curve of the Hamiltonian system defined by the function H , in which ξ(t) = ξ is defined by (4.5). The Hamiltonian system defined by the function H is the system of ordinary differential equations in the (x, ξ )-space, the phase space of classical mechanics, defined by the equations (4.7) and (4.8) below. In our case, 1 g(x)(v − b(x), v − b(x)), (4.6) 2 which yields g(x)(v − b(x)) = ξ or v = b(x) + a(x)ξ , and the formula (4.3) for H (x, ξ ) readily follows. It is proved in [2, Lemma 3.1, p. 120] that (4.2) holds for every t ∈ [0, T ], if γ is a minimizing curve. Because the substitution of ξ = g(x)(v − b(x)) and (4.6) in (4.3) yields that L(x, v) =

1 H = g(x)(v, v − b(x)) − g(x)(v − b(x), v − b(x)) 2 1 1 = g(x)(v, v) − g(x)(b(x), b(x)), 2 2 it follows that the condition (4.2) is equivalent to the condition that H ≡ 0 along the solution curves of the Hamiltonian system.

A well-known general property of the Legendre transform is that the function L can be found back from the function H by means of the formula L(x, v) = x, ξ − H (x, ξ ), where ξ = ξ(v) is the solution of the equation ∂H (x, ξ )/∂ξ = v. In our case we read


65

from (4.6) and g(x)(v − b(x)) = ξ , v − b(x) = a(x)ξ that L = a(x)(ξ, ξ )/2. Our recipe for minimizing curves therefore is to look among the solutions (x(t), ξ(t), s(t)) of the system of ordinary differential equations dxi /dt = ∂H (x, ξ )/∂ξi , dξi /dt = −∂H (x, ξ )/∂xi , ds/dt = a(x)(ξ, ξ )/2,

(4.7) (4.8) (4.9)

for those which satisfy x(0) = x, x(T ) = y, H (x(0), ξ(0)) = 0, s(0) = 0, and such that s(T ) is minimal. Note that H (x(0), ξ(0)) = 0 and (4.7) and (4.8) imply that H (x(t), ξ(t)) = 0 for every t. If x(t), 0 ≤ t ≤ T is a minimizing curve from x to y, then V (x, y) = s(T ). For a given point x ∈ M, the solutions of the Hamiltonian system which start at the points (x, ξ ) ∈ T∗ M such that H (x, ξ ) = 0 fill up a so-called Lagrange submanifold of the cotangent bundle T∗ M of M. This is a smoothly immersed n-dimensional submanifold of the 2n-dimensional phase space T∗ M such that the canonical two-form n dξi ∧ dxi i=1

of T∗ M vanishes identically on . If (x(t), ξ(t)) is a solution curve of the Hamiltonian system such that x(0) = x and H (x, ξ(0)) = 0, then for every T > 0 the curve x(t) with 0 ≤ t ≤ T is a candidate for being a minimizing curve from x to y = x(T ), and if this is the case, we have s(T ) = V (x, y). The s(T ) define a smooth function σ on the open subset + of which consists of the points (x(T ), ξ(T )) with T > 0. The projection from + to the base manifold M (the projection which forgets the ξ -components of the points of the phase space) is locally a diffeomorphism from an open neighborhood 0 in + of the point (y0 , η0 ) onto an open neighborhood M0 of y0 in M if and only if the tangent space of at the point (y0 , η0 ) is transversal to the tangent space of the fiber of the projection. If this is the case, then 0 can be written as the set of (y, η(y)) where y varies in M0 and η(y) depends smoothly on y ∈ M0 . In this case s(y) := σ (y, η(y)) defines a smooth function of y ∈ M0 . Moreover, η(y) = ds(y), which needs an argument. Proof. If γ (t) is a family of solutions of the Euler–Lagrange equations depending smoothly on the parameter , then in the variational equation only the boundary terms survive, viz. T ∂S ∂ ∂γ ∂L ∂γ ∂L = , , Ldt = − . ∂ ∂ 0 ∂ ∂v t=T ∂ ∂v t=0 (This is a classical observation of Hamilton.) If γ (0) = x for all , then the second term on the right-hand side is equal to zero, and recognizing ∂L/∂v as the momentum η(y), we arrive at v, ds(y) = v, η(y) if v = ∂γ (T )/∂ and y = γ (T ). On the other hand,

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∂ ∂T

0

T

∂γ ∂L , , = ∂t ∂v t=T

Ldt = L|t=T

in which the second equality follows from the condition that H = 0 along the corresponding solution curve of the Hamiltonian system; see (4.4) and (4.5). The tangent space of M at y = γ (T ) is spanned by the vectors ∂γ (T )/∂ and ∂γ (T )/∂T , where the γ (t) range over the arbitrary families of solutions of the Euler–Lagrange equations [L] = 0 with γ (0) = x and H = 0 along the corresponding solution of the Hamiltonian system. It follows that v, ds(y) = v, η(y) for every v ∈ Tv M, which means that ds(y) = η(y).

Because H = 0 on , it follows that the function s satisfies the nonlinear firstorder partial differential equation H (y, ds(y)) = 0. If the curves x(t) such that x(0) = x and x(T ) = y ∈ M0 are minimizing, then s(y) = V (x, y) and it follows that the function y → V (x, y) is smooth and satisfies the nonlinear first-order partial differential equation ∂V (x, y) H x, (4.10) = 0, y ∈ M0 . ∂y Moreover, the description in terms of s(y) leads to a quite explicit local construction of the function y → V (x, y). Remark 4.1. The partial differential equation (4.10) alone is far from sufficient to determine the function y → V (x, y) even if we add the condition that V (x, x) = 0. Remark 4.2. One can also look at the solutions (x(t), ξ(t)), −T ≤ t ≤ 0, of the Hamiltonian system on H = 0 such that x(0) = y, i.e., x(t) ends up at the given point y ∈ M. Here T > 0 and we have shifted the interval [0, T ] to [−T , 0] in order to have a fixed final time and a variable initial time (equal to −T ). Under conditions analogous to the conditions leading to (4.10), we have that ∂V (x, y) H x, − (4.11) = 0, x ∈ M0 , ∂x which is the same nonlinear first-order partial differential equation as (4.10), but with the vector field b(x) replaced by −b(x); see (4.3). If x is a hyperbolic equilibrium point of the unperturbed deterministic system dx/dt = b(x), then the Lagrange manifold has to be replaced by the unstable manifold of the equilibrium point (x, 0) of the Hamiltonian system. Here we note that it is a general fact that the unstable manifold of a hyperbolic equilibrium point of a Hamiltonian system is a Lagrange submanifold of the phase space. We also note that in this case the curve (x(t), ξ(t)) with 0 ≤ t ≤ T is replaced by a curve (x(t), ξ(t)) with −∞ < t ≤ T , and the conditions x(0) = x, H (x(0), ξ(0)) = 0 are replaced by the conditions that x(t) → x and ξ(t) → 0 as t → −∞. The quantity s(T ), which is the candidate for the value of V (x, y), has to be replaced by the limit of s(T ) − s(t) as t → −∞. Under conditions as in the text preceding (4.10), the function y → V (x, y)


67

locally satisfies the nonlinear first-order partial differential equation (4.10) even if x is an equilibrium point of the unperturbed deterministic system. In a similar way, if y is a hyperbolic equilibrium point of the unperturbed deterministic system, then the Lagrange manifold is replaced by the stable manifold of the equilibrium point (y, 0) of the Hamiltonian system, the curve (x(t), ξ(t)) with 0 ≤ t ≤ T is replaced by a curve x(t), ξ(t)) with 0 ≤ t < ∞, and the condition that x(T ) = y is replaced by the conditions that x(t) → y and ξ(t) → 0 as t → ∞. Furthermore, the quantity s(T ), which is the candidate for the value of V (x, y), has to be replaced by the limit of s(t) as t → ∞. Under the natural geometric conditions discussed before, the function x → V (x, y) locally satisfies the nonlinear first-order partial differential equation (4.11) even if y is an equilibrium point of the unperturbed deterministic system. In general, there may exist x, y ∈ M for which no minimizing curves exist between x and y even if we allow the aforementioned curves which run in infinite time from and to the equilibrium point x and y, respectively. One cause can be that the minimum is attained by a chain of stationary curves from x to y, which runs via a sequence of equilibrium points of the unperturbed deterministic system. It could also happen that the infimum is approached by a sequence of curves which run out of a sequence of compact subsets of M which absorbs M. Often, as in our models for geomagnetic reversals, one assumes conditions which imply that the latter does not occur. Even if minimizing curves exist, it can happen that the Lagrange manifold + is constituted in such a way that for y in a neighborhood of y0 there is a number of different η = η(j ) (y), depending smoothly on y, such that (y, η(j ) (y)) ∈ + , leading to different competing candidates sj (y) = σ (y, η(j ) (y)) for the function y → V (x, y), which is equal to the minimum over j of the functions sj . Let Mj denote the region where V (x, y) is equal to the smooth function sj (y).At the transition between the region Mj and Mk with k = j , the function y → V (x, y) is still continuous, but only piecewise smooth instead of smooth. Such boundaries between the region Mj resemble phase transitions in statistical mechanics. Also the functions sj (y) themselves can develop singularities, for instance, when (y, dsj (y)) approaches points at which is no longer transversal to the fiber of the projection onto the base manifold. This phenomenon is analogous to the occurrence of caustics in geometrical optics. This description of the minimizing curves in terms of the Hamiltonian system is not mentioned in [10] and [2]. It is an example of the application of symplectic geometry to variational calculus, and via Freidlin–Wentzell theory to stochastic perturbations of dynamical systems.

5 Hoyng’s model Hoyng’s model for the earth’s magnetic field is a stochastic perturbation of a deterministic system which has two stable equilibria (corresponding to the present average magnetic field and its opposite), of which the domains of attraction are separated by

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the stable manifold of a saddle point at the origin (corresponding to the zero magnetic field). Another important feature of his model is that the stochastic vector fields are linear. Therefore also the stochastic fluctuations vanish at the origin, and the stochastic process which starts at the origin will remain there with probability one. One of the problems in the theory is to obtain estimates which ensure that the process which gets close to the origin will not remain there for too long a time in such a way that we may consider the origin as stochastically isolated from the complement of the origin. If this holds, then we can take as our configuration space M the complement of the origin in the vector space. (The elements of the vector space V represent the magnetic fields of the earth.) A heuristic argument that the origin is stochastically isolated from the complement of the origin is that if we replace the unperturbed deterministic vector field b(x) by its linear approximation b (o)x at the origin o, then the stochastic differential equation is invariant under the homotheties x → cx for any c > 0. It follows that if we parametrize the complement of the origin by x = es u, in which s ∈ R and u is a point on the unit sphere U , then we obtain a stochastic differential equation on R × U which is invariant under the translations (s, u) → (s +a, u), a ∈ R. Such a stochastic differential equation is complete in the sense that it has a well-defined stochastic process for all positive times, and the completeness for s → −∞ corresponds to the stochastic isolation of the origin in V from the complement M ! R × U of the origin in V . Because the configuration space M is not compact and the domain of attraction of a stable equilibrium point s of b(x) is not relatively compact, we cannot apply the theory of [10], [2] directly to our situation. However, we believe that the arguments can be extended to prove the analogous statements. In particular we think that as a consequence of the fact that the boundary of is equal to the stable manifold of the saddle point at the origin o, the most probable way of leaving one of the domains of attraction is via a neighborhood of o. This corresponds to a heteroclinic connection from the hyperbolic equilibrium point (s, 0) to the equilibrium point (o, 0) of the Hamiltonian system. Moreover, we conjecture that the mean time of exit is asymptotically equal to 2 2 V (s,o)/ e , modulo factors eη/ with arbitrarily small |η|. Here it may be instructive to observe that if we replace the unperturbed deterministic vector field b(x) by its linearization b (o)x at the origin, then the invariance of the stochastic differential equation under homotethies implies that V (cx, o) = V (x, o) for every x ∈ V and every c > 0, which means that the function V (x, o) only depends on the direction of the vector x and not on its distance to the origin. Because V (x, o) = 0 when x belongs to the stable manifold of the origin and the function x → V (x, o) is not identically equal to zero, this implies that the function x → V (x, o) is not continuous at the origin o. We conjecture that such a discontinuous behavior of the function x → V (x, o) at the origin is inherited by any vector fields and the deterministic vector field vanishes at the origin. This discontinuity is analogous to the discontinuity at the origin of the mean exit time, which was mentioned in the introduction.


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6 A very simple prototype For the unperturbed deterministic system, we take the system x˙ = x(1 − x 2 ),

y˙ = −2y

in the (x, y)-plane, which has stable equilibria at (1, 0) and (−1, 0), with domains of attraction equal to the right and left half-plane, respectively. The origin (0, 0) is an equilibrium point of saddle point type. Its stable manifold is equal to the y-axis, the common boundary of the two domains of attraction of the stable equilibrium points. (See Figure 1.) For the stochastic vector fields, we take x∂/∂x, y∂/∂y, x∂/∂y, y∂/∂x, which leads to the Hamiltonian function H = x(1 − x 2 )p − 2yq + (x 2 + y 2 )(p 2 + q 2 )/2. Figure 2 shows the projections γ on the configuration space (the (x, y)-plane) of the solutions on the unstable manifold of the point ((x, y), (p, q)) = ((1, 0), (0, 0)). Note that the minimizing curves starting from the stable equilibrium point (1, 0) are parts of these curves γ . In order to see more clearly what happens with these curves near the origin, we show an enlargement there in Figure 3. An interesting feature of this picture is the appearance of caustics. Using symmetry arguments, one obtains that the minimizing curves are parts of the curves γ which are stopped at the x- and the y-axis. This leads to a much “quieter’’ picture, but still with a caustic near the origin. There is a curve C inside caustic with its end point at the cusp, which is the boundary between the region where s1 (x, y) < s2 (x, y) and V ((1, 0), (x, y)) = s1 (x, y) and the region where s2 (x, y) < s1 (x, y) and V ((1, 0), (x, y)) = s2 (x, y), where s1 (x, y) and s2 (x, y) are two competing smooth functions of (x, y) as described in Section 4. Correspondingly, the function (x, y) → V ((1, 0), (x, y)) is continuous, but has a jump in its gradient along the curve C. Note that in the notation the points x and y in M in Section 4 have been replaced by (1, 0) and (x, y), respectively. The necessity of competing minimal curves can be explained as a consequence of the fact that S(γ ) = ∞ if γ runs on the x-axis from (1, 0) to (0, 0). This implies that the minimizing curve from (1, 0) to (x, 0) with small positive x must make a detour in the upper or lower half-plane. On the other hand, if x is close to 1, the minimizing curve from (1, 0) to (x, 0) runs over the x-axis. The transition appears in the region where the minimizing curves which run along the x-axis compete with the minimizing curves which make a detour. (See Figure 4.) Figure 5 shows the most probable exit paths, both from the right half-plane and from the left half-plane. These exit via the origin. It can be proved that they not only have to make a detour in the upper and lower half-plane, but actually approach the origin tangentially to the y-axis, the stable manifold of the saddle point at the origin. In the higher-dimensional model, they generically approach the saddle point from the direction of the eigenvector of the linearized deterministic system corresponding to the negative eigenvalue which is closest to zero.

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Just for fun, Figure 6 shows the projections on the configuration space on the unstable manifold of the point ((1, 0), (0, 0)) if we take only x∂/∂y and y∂/∂x as the stochastic vector fields. In this case the Hamiltonian function is equal to

H = x 1 − x 2 p − 2yq + x 2 q 2 + y 2 p 2 /2. Actually, this was the first toy example which Peter Hoyng gave me. The figure eights straddling the x-axis correspond to solutions of the Hamiltonian system which run to infinity in a finite time, while their projections in the configuration space converge to a limit point on the x-axis, running faster and faster through an infinite sequence of decreasing figure eights.

References [1] K. D. Elworthy, Stochastic Differential Equations on Manifolds, Cambridge University Press, London, 1982. [2] M. I. Freidlin and A. D. Wentzell, Random Perturbations of Dynamical Systems, SpringerVerlag, New York, 1998. [3] R. Z. Has’minskiˇı (Khas’minskii), Stochastic Stability of Differential Equations, Sijthoff and Noordhoff, Alphen aan den Rijn, The Netherlands, 1980. [4] P. Hoyng, M.A. J. H. Ossendrijver, and D. Schmitt, The geodynamo as a bistable oscillator, Geophys. Astrophys. Fluid Dynam., 94 (2001), 263–314. [5] P. Hoyng, D. Schmitt, and M. A. J. H. Ossendrijver, A theoretical analysis of the observed variablity of the geomagnetic dipole field, Phys. Earth Planetary Interiors, 130 (2002), 143–157. [6] N. Ikeda and S. Watanabe: Stochastic Differential Equations and Diffusion Processes, North-Holland, Amsterdam, 1981. [7] R. T. Merrill, M. W. McElhinny, and P. L. McFadden, The Magnetic Field of the Earth, Academic Press, New York, 1966. [8] B. Øksendal, Stochastic Differential Equations, 1st ed., Springer-Verlag, Berlin, 1989; 5th ed., 1998. [9] M. A. J. H. Ossendrijver, P. Hoyng, and D. Schmitt, Stochastic excitation and memory of the solar dynamo, Astron. Astrophys., 313 (1996), 938–948. [10] A. D. Wentzell and M. I. Freidlin, On small random perturbations of dynamical systems, Russian Math. Surveys, 25-1 (1970), 1–55.

Nonholonomic systems via moving frames: Cartan equivalence and Chaplygin Hamiltonization∗ Kurt Ehlers1 , Jair Koiller2 , Richard Montgomery3 , and Pedro M. Rios4 1 Department of Mathematics

Truckee Meadows Community College 7000 Dandini Boulevard Reno, NV 89512-3999 USA [email protected] 2 Fundação Getulio Vargas Praia de Botafogo 190, Rio de Janeiro 22253-900 Brazil [email protected] 3 Mathematics Department University of California at Santa Cruz Santa Cruz, CA 95064 USA [email protected] 4 Department of Mathematics University of California at Berkeley Berkeley, CA 94720 USA [email protected] Dedicated to Alan Weinstein on his 60th birthday. Abstract. A nonholonomic system, for short “NH,’’ consists of a configuration space Qn , a Lagrangian L(q, q, ˙ t), a nonintegrable constraint distribution H ⊂ T Q, with dynamics governed by Lagrange–d’Alembert’s principle. We present here two studies, both using adapted moving frames. In the first we explore the affine connection viewpoint. For natural Lagrangians L = T −V , where we take V = 0 for simplicity, NH-trajectories are geodesics of a (nonmetric) connection ∇N H which mimics Levi-Civita’s. Local geometric invariants are obtained by Cartan’s method of equivalence. As an example, we analyze Engel’s (2–4) distribution. This is the first such study for a distribution that is not strongly nonholonomic. In the second part we study ∗ The authors thank the Brazilian funding agencies CNPq and FAPERJ: a CNPq research

fellowship (JK), a CNPq post-doctoral fellowship at Berkeley (PMR), a FAPERJ visiting fellowship to Rio de Janeiro (KE). (JK) thanks the E. Schrödinger Institute, Vienna, for financial support during Alanfest and the Poisson Geometry Program, August 2003.

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K. Ehlers, J. Koiller, R. Montgomery, and P. M. Rios

G-Chaplygin systems; for those, the constraints are given by a connection φ : T Q → Lie(G) on a principal bundle G → Q → S = Q/G and the Lagrangian L is G-equivariant. These systems compress to an almost Hamiltonian system (T ∗ S, H φ , N H ), N H = can +(J.K), with d(J.K) = 0 in general; the momentum map J : T ∗ Q → Lie(G) and the curvature form K : T Q → Lie(G)∗ are matched via the Legendre transform. Under an s ∈ S dependent time reparametrization, a number of compressed systems become Hamiltonian, i.e., N H is sometimes conformally symplectic. A necessary condition is the existence of an invariant volume for the original system. Its density produces a candidate for conformal factor. Assuming an invariant volume, we describe the obstruction to Hamiltonization. An example of a Hamiltonizable system is the “rubber’’ Chaplygin’s sphere, which extends Veselova’s system in T ∗ SO(3). This is a ball with unequal inertia coefficients rolling without slipping on the plane, with vertical rotations forbidden. Finally, we discuss reduction of internal symmetries. Chaplygin’s “marble,’’ where vertical rotations are allowed, is not Hamiltonizable at the compressed T ∗ SO(3) level. We conjecture that it is also not Hamiltonizable when reduced to T ∗ S 2 . “Nonholonomic mechanical systems (such as systems with rolling contraints) provide a very interesting class of systems where the reduction procedure has to be modified. In fact this provides a class of systems that give rise to an almost Poisson structure, i.e., a bracket which does not necessarily satisfy the Jacobi identity’’ (Marsden and Weinstein [2001]).

1 Introduction and outline Cartan’s moving frames method is a standard tool in Riemannian geometry.1 In analytical mechanics, the method goes back to Poincaré [1901], perhaps earlier, to Euler’s rigid body equations, perhaps much earlier, to the cave person who invented the wheel. Let q ∈ Rn be local coordinates on a configuration space Qn , and consider a local frame, defined by an n × n invertible matrix B(q), ∂ ∂ = bij , ∂πj ∂qi

n

Xj =

π˙ j Xj =

i=1

q˙i

∂ , ∂qi

π˙ = A(q)q, ˙

A = B −1 .

(1.1) In mechanical engineering (Hamel [1949], Papastavridis [2002]), moving frames are disguised under the keyword quasi-coordinates, nonexisting entities π such that ∂f ∂qi ∂f ∂f = = bij = Xj (f ). ∂πj ∂qi ∂πj ∂qi i

i

Let {i }i=1,...,n be the dual coframe to {Xj }, i = “dπi ’’ =

j

aij dqj .

1 Cartan [1926]; there is a recent English translation from the Russian translation (Cartan

[2001]). One of the most important applications was the construction of characteristic classes by Alan’s advisor, S. S. Chern. Our taste for moving frames in mechanics is a small tribute to his influence.

Nonholonomic systems via moving frames

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1.1 Moving frames: Lagrangian and Hamiltonian mechanics The Euler–Lagrange 1-form may be rewritten as:2 n ∂L d ∂L − − Fr dqr dt ∂ q˙r ∂qr r=1 ⎛ ⎞ n n n ∗ ∗ ∗ ∂L ∂L d ∂L ⎝ = − + γkji π˙ j − Rk ⎠ k = 0, dt ∂ π˙ k ∂πk ∂ π˙ i k=1

i=1

(1.2)

j =1

where L∗ (q, π˙ , t)= L(q, B(q)π˙ , t) is the Lagrangian written in “quasi-coordinates’’ and Rk = s Fs bsk are the covariant components of the total force (external, Fext , and constraint force λ). The so-called Hamel transpositional symbols γkji = γjik = ns,=1 bsk bj (∂ais /∂q − ∂ai /∂qs ) are precisely the moving frame structure coefficients (Koiller [1992]). If the velocities are restricted to a subbundle H ⊂ T Q, a constraint force λ appears. The d’Alembert–Lagrange principle3 implies that λ belongs to the anihilator Ho ⊂ T ∗ Q of H, hence exerting zero work on admissible motions q˙ ∈ H: [L] :=

d ∂L ∂L − − Fext = λ ∈ Ho , dt ∂ q˙ ∂q

q˙ ∈ H.

(1.3)

Using moving frames, constraints can be eliminated directly. If Ho is spanned by the last r forms J , s + 1 ≤ J ≤ n (s = n − r), then equations of motion result from setting the first s Euler–Lagrange differentials equal to zero: n n d ∂L∗ ∂L∗ ∂L∗ i − + γkj π˙ j − Fkext = 0 dt ∂ π˙ k ∂πk ∂ π˙ i i=1

(1 ≤ k ≤ s).

(1.4)

j =1

Strikingly, the Hamiltonian counterparts of (1.2) and (1.4) are simpler, although terms of the less known.4 The philosophy is to fight against Darboux’s dictatorship. In local coframe {i }1≤i≤n , any element pq ∈ T ∗ Q can be written as pq = mi i (q). The natural 1-form α on T ∗ Q keeps the familiar confusing expression α := pdq = m. Consequently, the canonical symplectic form := dα may be written as

:= dp ∧ dq = dm ∧ + md.

(1.5)

The second term md, which deviates from Darboux’s format, is not a nuisance; it carries most valuable information. For instance, Kostant–Arnold–Kirillov–Souriau’s bracket in T ∗ G, G a Lie group, can be immediately visualized: take a (left- or right-) 2 Atributed to Hamel, but certainly known by Poincaré. Quasi-coordinates can be found in

Whittaker [1937] and were first used in mechanics by Gibbs; see Pars [1965]. 3 According to Sommerfeld [1952], this gives the most natural foundation for mechanics.

4 A “moving frames operational system’’ for Hamiltonian mechanics in T ∗ Q was given in

Koiller, Rios, and Ehlers [2002].

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invariant coframe and apply H. Cartan’s “magic formula’’ on d. So moving frames are ideally suited when a Lie symmetry group G is present.5 Example: Mechanics in SO(3) To fix notation, we now review the standard example. The Lie algebra basis Xi ∈ sO(3) = TI SO(3), i = 1, 2, 3 (infinitesimal rotations around the x, y, z-axis at the identity) can either be right or left transported, producing moving frames on SO(3) denoted {Xir } and {Xi }, respectively. Let {ρi }1≤i≤3 and {λi }1≤i≤3 denote their dual coframes (right- and left-invariant forms in SO(3)). To represent angular momenta, we use Arnold’s notations (Arnold [1989]): capital letters mean objects in the body frame, lowercase objects in the space frame. Thus for instance, = RL, where L is the angular momentum in the body frame and is the angular momentum in space; likewise ω = R relate the angular velocities. The canonical 1-form in T ∗ SO(3) is given by α = 1 ρ1 + 2 ρ2 + 3 ρ3 = L1 λ1 + L2 λ2 + L3 λ3 , so

can = =

di ρi + 1 dρ1 + 2 dρ2 + 3 dρ3 dLi λi + L1 dλ1 + L2 dλ2 + L3 dλ3 ,

where by Cartan’s structure equations, dλ1 = −λ2 ∧ λ3 , . . . and dρ1 = ρ2 ∧ ρ3 , . . . (cyclic). A left-invariant metric is given by an inertia operator L = A . Euler’s rigid body equations follow immediately. Poisson action of S 1 on SO(3) Consider the left S 1 action on SO(3) given by exp(iφ) · R := S(φ)R, where S(φ) is the rotation matrix about the z-axis: ⎛ ⎞ ⎛ ⎞ cos(φ) − sin(φ) 0 0 −1 0 S(−φ)S (φ) = ⎝ 1 0 0 ⎠ = X3 . S(φ) := ⎝ sin(φ) cos(φ) 0 ⎠ , 0 0 1 00 0 Two matrices are in the same equivalence class iff their third rows, which we denote by γ , called the Poisson vector, are the same: R1 ∼ R2 ⇐⇒ R1−1 kˆ = R2−1 kˆ = γ ∈ S 2 . ˆ The So we have a principal bundle π : SO(3) → S 2 , γ = π(R) = R −1 kˆ = R † k. derivative of π is −1 ˙ = −(R −1 RR ˙ −1 )k = −(R −1 R)(R ˙ γ˙ = π∗ (R) )k = −[ ]γ = − × γ = γ × , (1.6) 5 As we learned from Alan at the banquet, the etymology for symplectic is “capable to join,’’

themes and people. The latter is one of the most important aspects of the symplectic “creed.’’ Provocation: taking moving frames, adapted to some other mathematical structure for Q, would the non-Darboux term provide a local symplectic invariant?


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where we used the customary identification6 [ ] ∈ sO(3) ↔ ∈ R3 , Arnold [1989]. The lifted action to T ∗ SO(3) has momentum map J = 3 . Connection on S 1 → SO(3) → S 2 Take the usual bi-invariant metric , on SO(3) so that both {Xi } and {Xir } are orthonormal moving frames. The tangent vectors to the fibers are (d/dφ)S(φ) · R = right X3 . Consider the mechanical connection associated to , , namely, that horizonright tal and vertical spaces are orthogonal. The horizontal spaces are generated by X1 right and X2 . The connection form is φ = ρ3 . The horizontal lift of γ˙ to R is the tangent vector R˙ such that (1.7)

hor = R −1 R˙ = [γ˙ × γ ]. Note that hor is the −90 degrees rotation of γ˙ inside Tγ S 2 . The curvature of this connection κ = dρ3 is the area form of the sphere. Reduction of S 1 symmetry It is convenient for reduction to use (a, 3 ), a ∈ R3 , a ⊥ γ , L := a × γ + 3 γ ,

(1.8)

where a is a vector perpendicular to γ . The vector a has an intrinsic meaning: Consider a moving frame e1 , e2 in S 2 , with dual coframe θ1 , θ2 . Then vγ = v1 e1 + v2 e2 parametrizes T S 2 , and pγ = a · dγ = p1 θ1 + p2 θ2 parametrizes T ∗ S 2 , a = γi dγi = 0 denotes both an element of T ∗ S 2 and the p1 e1 + p2 e2 . Here a · dγ , canonical 1-form. Our parametrization for SO(3) is R(φ, γ ) = S(φ) · R(γ ), R(γ ) = rows(e1 , e2 , γ ). Then L = p2 e1 − p1 e2 + 3 γ corresponds to = (p2 , −p1 , 3 ) along the section φ = 0. The right-invariant forms are compactly represented as ρ3 = dφ − (de1 , e2 ),

ρ1 + iρ2 = −i exp(iφ)(θ1 + iθ2 ).

(1.9)

Lifting v ∈ T S 2 to an horizontal vector in T SO(3) is simple:

hor = [(v1 e1 + v2 e2 ) × γ ] = [v2 e1 − v1 e2 ] or

hor(v) = v2 X1r − v1 X2r . (1.10)

Hence any vector R˙ ∈ T SO(3) can be written as R˙ = ω1 X1 + ω2 X2 + ω3 X3 with ω1 = v2 , ω2 = −v1 . Any covector pR ∈ T ∗ SO(3) can be written as pR = p1 π ∗ (θ1 ) + p2 π ∗ (θ2 ) + 3 ρ3 . The reduced symplectic manifold J −1 (3 )/S 1 ≡ T ∗ S 2 can be explicitly constructed, taking the section φ = 0. Let i : T ∗ S 2 → T ∗ SO(3), i(γ , p1 , p2 ) = (R(γ ), ),

= (p2 , −p1 , 3 ).

(1.11)

6 We will drop the [•] and • in what follows and mix all notation, hoping no confusion will arise. Equation (1.6) is one half of every system of ODEs for S 1 -equivariant mechanics in

SO(3). Of course, we also obtain γ˙ = − × γ by differentiating Rγ = k (we could use the notation γ = K, but we won’t).

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Then from (1.9) we get i ∗ ρ2 = −θ1 , i ∗ ρ1 = θ2 , and i ∗ d = di ∗ yields i ∗ dρ1 = dθ2 ,

i ∗ dρ2 = −dθ1 ,

i ∗ dρ3 = i ∗ ρ1 ∧ i ∗ ρ2 = −θ2 θ1 = θ1 θ2 .

We get immediately

red = i ∗ ( T ∗ SO(3) ) = d(p1 θ1 + p2 θ2 ) + 3 area = can + 3 areaS2 . (1.12) T ∗S2 T ∗S2 All references to the moving frame disappear, but the expression can = d(p1 θ1 + T ∗S2 p2 θ2 ) suggests that whenever a natural mechanical system in T ∗ SO(3) reduces to T ∗ S 2 ≡ T S 2 , there is a preferred choice for the moving frame {e1 , e2 }γ : namely, that which diagonalizes the Legendre transform Tγ S 2 → Tγ∗ S 2 ≡ Tγ S 2 of the reduced (Routh) Lagrangian. 1.2 Nonholonomic systems A NH system (Q, L, H) consists of a configuration space Qn , a Lagrangian L : T Q × R → R, and a totally nonholonomic constraint distribution H ⊂ T Q. The dynamics are governed by Lagrange–d’Alembert’s principle.7 Usually L is natural, L = T − V , where T is the kinetic energy associated to a Riemannian metric , , and V = V (q) is a potential. By totally nonholonomic, we mean that the filtration H ⊂ H1 ⊂ H2 ⊂ · · · ends in T Q. Each subbundle Hi+1 is obtained from the previous one by adding to Hi combinations of all possible Lie brackets of vector fields in Hi . To avoid interesting complications we assume that all have constant rank. Equivalently, let Ho ⊂ T ∗ Q the codistribution of “admissible constraints’’ annihilating H; dually, one has a decreasing filtration of derived ideals ending in zero. Internal symmetries of NH systems: Noether’s theorem An internal symmetry occurs whenever a vector field ξQ ∈ H preserves the Lagrangian. For natural systems ξQ is a Killing vector field for the metric. Noether’s theorem from unconstrained mechanics remains true. The argument (see Arnold, Kozlov, and Neishtadt [1988]) goes as follows: denote by φξ (s) the one-parameter d group generated by ξ and let φ(s, t) = φξ (s) · q(t), so φ = ds φ = ξQ (φ), where q(t) is chosen as a trajectory of the nonholonomic system. Differentiating with red spect to s the identitly L(φ(s, t), dt φ(s, t)) = const after a standard integration by d ∂L parts we get dt ( ∂ q˙ φ ) = [L]φ . This vanishes precisely when φ = ξQ ∈ H, so Iξ :=

∂L ∂ q˙

· ξ = const.

7 “Vakonomic’’ mechanics uses the same ingredients, but the dynamics are governed by the

variational principle with constraints, and produce different equations; see, e.g., Cortés, de Léon, de Diego, and Martínez [2003]. The equations coincide if and only if the distribution is integrable. In spite of many similarities, there are striking differences between NH and holonomic systems. For instance, NH systems do not have (in general) a smooth invariant measure. Necessary and sufficient conditions for the existence of the invariant measure were first given (explicitly in coordinates) by Blackall [1941].


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External symmetries: G-Chaplygin systems External (or transversal) symmetries occur when group G acts on Q, preserving the Lagrangian and the distribution H, meaning that g∗ Hq = Hgq . In the most favorable case one has a principal bundle action Gr → Qn → S m , m + r = n, where H forms the horizontal spaces of a connection with 1-form φ : T Q → Lie(G). These systems are called G-Chaplygin.8 Terminology ´ Since Bates and Sniatycki [1993], and Bloch, Krishnaprasad, Marsden, and Murray [1996], several authors have called attention to these two types of symmetries. Re´ duction of internal symmetries was already described in Sniatycki [1998]. To stress the difference, reduction of external symmetries is called compression here. The word reduction will be used for internal symmetries. LR systems Veselov and Veselova [1986], Veselov and Veselova [1988] considered Lie groups Q = G with left-invariant metrics, with constraint distributions given by right translation of D ⊂ Lie(G), i.e., the constraints are given by right-invariant forms. For a LR-Chaplygin system, in addition there is a decomposition Lie(G) = Lie(H ) ⊕ D, where H is a Lie subgroup such that Ad h−1 D = h−1 Dh = D. Therefore, H → G → S = G/H is a H -Chaplygin system; the base S is the homogeneous space of cosets H g. Fedorov and Jovanovic [2003] considered the case where G is compact and Lie(H ) is orthogonal to D with respect to the bi-invariant metric.9 Compression of G-Chaplygin systems From symmetry, it is clear that the Lagrange–d’Alembert equations compress to the base T S.10 In covariant form, the dynamics take the form [Lφ ] = F (s, s˙ ), where Lφ (s, s˙ ) = L(s, h(˙s )) is the compressed Lagrangian in T S; h(˙s ) is the horizontal 8 A“historical’’remark (by JK). Chaplygin considered the abelian case. During a post-doctoral

year in Berkeley, way back in 1982, I became interested in NH systems with symmetries. Alan directed me to two wonderful books: Hertz [1899] Foundation of Mechanics and Neimark and Fufaev [1972]. In the latter I learned about (abelian) Chaplygin systems, presented in coordinates. I said to Alan that I would like to examine nonabelian group symmetries, and Alan immediately made a diagram on his blackboard, and told me: “well, then, the constraints are given by a connection on a principal bundle.’’ This was the starting point of Koiller [1992]. 9 These conditions are not met in the marble and rubber Chaplygin spheres (see Section 3.2); however, Veselov’s result (Theorem 3.3 below) on invariant volume forms still holds. 10 The full dynamics can be reconstructed from the compressed solutions, horizontal lifting the trajectories via φ, since the admissible paths are horizontal relative to the connection. This last step is not “just’’ a quadrature; in the nonabelian case, a path-ordered integral is in order. For G = SO(3), Levi [1996] found an interesting geometric construction.

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lift to any local section and F is a pseudogyroscopic force.11 In order to write F explicitly, take group quasi-coordinates (s, s˙ , g, π˙ ). Write q = gσ (s), with g ∈ G and a local section σ (s) of Q → S. Fix a basis Xk for the Lie algebra, [XK , XL ] = J X , X(π cKL ˙) = π˙ I XI . Any tangent vector q˙ ∈ Tσ (s) Q can be written as J ˙ ))·σ (s). Horizontal vectors are represented by π˙ = b(s)·˙s , where q˙ = dσ (s)·˙s +X((π b(s) is an r ×m matrix. The connection 1-form may be written as φ(q) ˙ = π˙ −b(s)· s˙ . Then ⎛ ⎞ ∗ m r r b ∂L b K ⎠ ⎝ Ki − Kj + [Lφ ] = F (s, s˙ ), F = s˙j . bU i bVj cU V ∂ π˙ k ∂qj ∂qi K=1

j =1

U,V =1

(1.13) 1.3 Main results Using the moving frames method we present results on two aspects of nonholonomic systems. • •

Cartan’s equivalence, using Cartan’s geometric description of NH systems via affine connections (Cartan [1928]). The objective is to find all local invariants. Chaplygin systems: compression of external symmetries, reduction of internal symmetries. The objective is to generalize Chaplygin’s “reducing factor’’ method (Chaplygin [1911]), namely, verify if Hamiltonization is possible (via conformally symplectic structures).

Results on Cartan’s equivalence In Section 2 we analyze NH systems under the affine connection perspective. We pursue the (local) classification program proposed by Cartan [1928] using his equivalence method. See Koiller, Rodrigues, and Pitanga [2001] and Tavares [2002] for a rewrite of Cartan’s paper in modern language. Cartan’s method of equivalence is a powerful method for uncovering and interpreting all differential invariants and symmetries in a given geometric structure. In Ehlers [2002] NH systems in a 3-manifold with a contact distribution were classified. Here we go one step further, looking at Engel’s distribution in 4-manifolds (see definition below). Our results are summarized in Theorem 2.3. The “role model’’ here is the rolling penny example (no pun intended). This is the first such study for a distribution that is not strongly nonholonomic. Next in line is studying the famous Cartan 2–3–5 distribution. Results on G-Chaplygin systems Instead of using (1.13) in TS, we may describe the compressed system in T ∗ S as an 11 This nonholonomic force represents, philosophically, a concealed force in the sense of Hertz

[1899], having a geometric origin. This force vanishes in some special cases, not necessarily requiring the constraints to be holonomic. Equivalently, the dynamics in T S is the geodesic spray of a modified affine connection. One adds to the induced Levi-Civita connection in T S a certain tensor B(X, Y ). This NH connection in general is nonmetric (Koiller [1992]).


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almost Hamiltonian system12 iX N H = dH,

H = H φ : T ∗ S → R,

∗

T S

N H = can + (J.K),

(1.14)

where H φ is the Legendre transform of the compressed Lagrangian. (J.K) is a semibasic 2-form on T ∗ S which in general is not closed. As one may guess, J is the momentum map, and K is the curvature of the connection. Ambiguities cancel, since J is Ad ∗ -equivariant while K is Ad-equivariant. The construction is independent of the point q on the fiber over s. Under an s ∈ S dependent time reparametrization, dτ = f (s)dt, several interesting compressed G-Chaplygin systems become Hamiltonian. A necessary condition is the existence of an invariant volume (Theorem 3.3) whose density F produces a candidate f = F 1/(m−1) , m = dim(S) for a conformal factor. Chaplygin’s “rubber’’ ball (vertical rotations forbidden) is, as far we know, a new example, and generalizes the well-known Veselova system in SO(3) (Proposition 3.6). We describe the obstruction to Hamiltonization as the 2-form iX d(f N H ) (Theorem 3.4) and we discuss further reduction by internal symmetries. An example of the latter situation is Chaplygin’s “marble’’ (a hard ball with unequal inertia coefficients rolling without slipping on the plane). It is non-Hamiltonizable in T ∗ SO(3), and our calculations suggest that it is also non-Hamiltonizable when reduced to T ∗ S 2 (Theorem 3.8). Compare with Borisov and Mamaev [2001]. What does Hamiltonization accomplish? Why do we focus so much on the question of Hamiltonizability? The example of the reduced equations for Chaplygin’s skate (after a two-dimensional Euclidean symmetry is removed) shows that changing time scale in a nonholonomic systems can completely change its character. In this example (see, e.g., Koiller [1992]) the fully reduced equations of motion are not Hamiltonian because every solution is asymptotic in forward and backward time to a point which depends on which solution you choose. However, after rescaling time the fully reduced equations become Hamiltonian, namely, the harmonic oscillator. However, this Hamiltonian vector field is incomplete because along one of the coordinate axes, the time rescaling is not defined.13 In light of this example, why is time rescaling interesting? The answer is that it is interesting mostly in the context of integrability, where no singularities are removed in the phase space. See Section 3.

2 Nonholonomic geometry: Cartan equivalence A Cartan nonholonomic structure is a triple (Q, G = ·, ·, H), where Q is an ndimensional manifold endowed with a Riemannian metric G and a rank r totally 12 For details, see Koiller, Rios, and Ehlers [2002], Koiller and Rios [2001]. The Hamiltonian

compression for Chaplygin systems was first explored, in the abelian case, by Stanchenko [1985]. The nonclosed term was described as a semibasic 2-form, depending linearly on the fiber coordinate in T ∗ S, but its geometric content was not indicated there. 13 We thank one of the referees for this observation.

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nonholonomic distribution H. Our motivation for studying such a structure is a free particle moving in Q, nonholonomically constrained to H, with kinetic energy T = 12 ·, ·. The nonholonomic geodesic equations are obtained by computing accelerations using the Levi-Civita connection associated with G and orthogonally projecting the result onto H. The projected connection is called a nonholonomic connection (Lewis [1998]), and was introduced by Cartan [1928]. A distribution H is strongly nonholonomic if any basis of vector fields spanning H on U ⊂ Q, together with their Lie brackets, span the entire tangent space over U . The equivalence problem for nonholonomic geometry was revisited in Koiller, Rodrigues, and Pitanga [2001] and the generalization to arbitrary nonholonomic distributions was discussed. Engel manifolds provide the simplest example involving distributions that are not strongly nonholonomic.14 The main question we address is the following. Given two nonholonomic struc¯ H), ¯ is there a (local) diffeomorphism f : U ⊂ Q → ¯ G, tures (Q, G, H) and (Q, ¯ carrying nonholonomic geodesics in Q to nonholonomic geodesics in Q? ¯ U¯ ⊂ Q In Cartan’s approach, this question is recast as an equivalence problem. The nonholonomic structure is encoded into a subbundle of the frame bundle over Q called a G-structure. The diffeomorphism f exists if the two corresponding G-structures are locally equivalent. Necessary and sufficient conditions for the G-structures to be equivalent are given in terms of differential invariants found using the method of equivalence. Outline Our main example is the equivalence problem for nonholonomic geometry on an Engel manifold. Let Q be a four-dimensional manifold and H a rank two distribution. H is an Engel distribution if and only if, for any vector fields X and Y locally spanning H, and some functions a, b : Q → R, the vector fields X, Y , Z = [X, Y ], and W = a[X, Z] + b[Y, Z] form a local basis for T Q. By an Engel manifold, we mean a fourdimensional manifold endowed with an Engel distribution. We begin by describing the nonholonomic geodesic equations. In the spirit of Cartan’s program, we express them in terms of connection 1-forms and (co)frames adapted to the distribution. This formulation is particularly well suited to the problem at hand; the nonholonomic geodesic equations are obtained by writing the ordinary geodesic equations in terms of the Levi-Civita connection 1-form and crossing out terms corresponding to directions complementary to H. We then set up the equivalence problem for nonholonomic 14 Historical remarks. Cartan [1928] introduced the equivalence problem for nonholonomic

geometry and studied the case of manifolds endowed with strongly nonholonomic distributions. In his address, Cartan warned against attempts to study other cases because of the “plus compliqués’’ computations involved. In the meantime strides have been made in the equivalence method by Robert Gardner and his students that allow computations to be made at the Lie algebra level rather than at the group level (Gardner [1989]). This together with symbolic computation packages such as MathematicaTM make equivalence problems tractable in many important cases. See Gardner [1989], Bryant [1994], Montgomery [2002], Grossman [2000], Ehlers [2002], Hughen [1995], and Moseley [2001] for some applications.


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geometry and give a brief description of the equivalence method as it is applied to our main example. We conclude this section by applying the method of equivalence to the case of nonholonomic geometry on an Engel manifold. We derive all differential invariants associated with the nonholonomic structure and show that the symmetry group of such a structure has dimension at most four. 2.1 Nonholonomic geodesics: Straightest paths Totally nonholonomic distributions A distribution H is a rank r vector subbundle of the tangent bundle T (Q) over Q. Let H1 = H + [H, H] and Hi = [H, Hi ], and consider the filtration H ⊂ H1 ⊂ · · ·Hi ⊂ · · · ⊂ T Q. H is totally nonholonomic if and only if, for some k, Hk = T Q at all points in Q. For the present discussion we will assume that each Hi has constant rank over Q. As a specific example, consider the Engel distribution H on R4 with coordinates ∂ ∂ ∂ ∂ , X2 = ∂x + w ∂y + y ∂z }. There are, in fact, local (x, y, z, w), spanned by {X1 = ∂w coordinates on any Engel manifold so that the distribution is given by this normal form, see Montgomery [2002]. Then {X1 , X2 , X3 = [X1 , X2 ]} spans the three-dimensional distribution H1 , and {X1 , X2 , X3 , X4 = [X2 , X3 ]} spans the entire T R4 . A path c : R → Q is horizontal if c(t) ˙ ∈ Hc(t) for all t. Chow’s theorem implies that if H is totally nonholonomic, then any two points in Q can be joined by a horizontal path (see Montgomery [2002]). At the other extreme, the classical theorem of Frobenius implies that H is integrable, which is to say that Q is foliated by submanifolds whose tangent spaces coincide with H at each point, if and only if [Xi , Xj ] ∈ H for all i and j (Warner [1971]). In what follows we will need a description of distributions in terms of differential ideals. Details can be found in Warner [1971] or Montgomery [2002]. Let I = H⊥ be the ideal in ∗ (Q) consisting of the differential forms annihilating H. If H is rank r, then I is generated by n − r independent 1-forms. The first derived ideal of I is the ideal (I) := {θ ∈ I|dθ ≡ 0 mod(I)}. (2.1) If we set I (0) = I and I (n+1) = (I (n) ) we obtain a decreasing filtration I = I (0) ⊃ I (1) ⊃ · · · ⊃ 0. The filtration terminating with the 0 ideal is equivalent to the assumption that the distribution is completely nonholonomic. We note that I (j ) = (Hj )⊥ for j = 1, but this is not true in general for j > 1 (see Montgomery [2002]). At the other extreme, the differential ideal version of the Frobenius theorem implies that H is integrable if and only if (I) ⊂ I (Warner [1971]). For the Engel example, the 1-forms η1 = dy − wdx and η2 = dz − ydx generate the ideal I. Notice that dη2 = η1 ∧ dx so η2 ∈ I (1) but dη1 cannot be written in terms of η1 or η2 ; therefore, η1 ∈ / I (1) .

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The nonholonomic geodesic equations There are two different geometries commonly defined on a nonholonomic structure (Q, G = ·, ·, H): sub-Riemannian geometry and nonholonomic geometry. In sub-Riemannian geometry one is interested in shortest √ paths. The length of a path c : [a, b] → Q joining points x and y is (c) = c, ˙ cdt. ˙ The distance from x to y is d(x, y) = inf((c)) taken over all horizontal paths joining x to y. In nonholonomic geometry one is interested in straightest paths, which are solutions to the nonholonomic geodesic equations. Hertz [1899] was the first to notice that shortest = straightest unless the constraints are holonomic.15 The nonholonomic geodesic equations are obtained by computing the acceleration of a horizontal path c : R → Q using the Levi-Civita connection associated with G and orthogonally projecting the result onto H. It is convenient to adopt the following indicial conventions: 1 ≤ I, J, K ≤ n, 1 ≤ i, j, k ≤ r (= rank(H)), r + 1 ≤ ν ≤ n.

(2.2)

Let e = {eI } be a local orthonormal frame for which the ei span H, and let η = {ηI } be the dual coframe defined by ηI (eJ ) = δI J , the Kronecker delta function. We note that the ην annihilate H and the metric, restricted to H is g|H = η1 ⊗ η1 + · · · + ηr ⊗ ηr . The Levi-Civita connection can be expressed in terms of local 1-forms ωI J = −ωJ I satisfying Cartan’s structure equation dη = −ω ∧ η (Hicks [1965]). A horizontal path c : R → M is a nonholonomic geodesic if it satisfies the nonholonomic geodesic equations ⎡ ⎤ d ⎣ (vi ) + vj ωij (c) ˙ ⎦ ei = 0, (2.3) dt j

where 1 ≤ i, j, ≤ r and vi = ηi (c) ˙ are the quasi-velocities. Example: The vertical rolling penny Astandard example of a mechanical system modeled by a nonholonomic Engel system is that of a coin rolling without sliping on the Euclidean plane. Consider a coin of radius a rolling vertically on the xy-plane. The location of the coin is represented by the coordinates (x, y, θ, φ). The point of contact of the coin with the plane is (x, y), the angle made by the coin with respect to the positive x-axis is θ, and the angle made by the point of contact, the center of the coin, and a point marked on the outer edge of the coin is φ. The state space can be identified with the Lie group SE(2) × SO(2) where the first factor is the group of Euclidean motions locally parametrized by x, 15 The terminology straightest path for a nonholonomic geodesic was, in fact, coined by Hertz

himself.


87

y and θ. The mass of the coin is m, the moment of inertia in the θ direction is J and the moment of inertia in the φ direction is I . The kinetic energy, which defines a Riemannian metric on the state space, is T =

J I m (dx ⊗ dx + dy ⊗ dy) + dθ ⊗ dθ + dφ ⊗ dφ. 2 2 2

(2.4)

The penny rolls without slipping giving rise to the constraints ˙ x˙ = (a cos θ )φ,

˙ y˙ = (a sin θ )φ.

Consider the orthonormal frame (X1 , X2 , X3 , X4 ), where # ∂ ∂ ∂ 2 X1 := + a sin θ + a cos θ , ∂x ∂y dφ ma 2 + I # 2 ∂ , X2 := J ∂θ # ∂ 2 ∂ X3 := + cos θ − sin θ , m ∂x ∂y # ∂ 2 ∂ X4 := + sin θ cos θ . m ∂x ∂y

(2.5)

(2.6)

Note that the constraint subspace is H = span{X1 , X2 }, and H(1) = span{X1 , X2 , X3 }. The dual coframe is (η1 , η2 , η3 , η4 ), where $ # ma 2 + I J 1 2 dφ, η := dθ, η := 2 2 # # m m 3 4 (− sin θ dx + cos θ dy), η := (cos θ dx + sin θ dy − dφ). η := 2 2 (2.7) To compute the Levi-Civita connection form, we determine ω = [ωI J ] such that ωI J = −ωJ I and dη = −ω ∧ η. Using simple linear algebra, we find % % ⎛ ⎞ m m 3 √1 2 √1 η η 0 0 2 2 2 J (ma +I ) 2 J (ma +I ) ⎜ ⎟ ⎜ ⎟ ⎜ ⎟ % % ⎜ − √1 ⎟ m 1 m 3 1 √ η 0 − η 0 ⎜ ⎟ 2 J (ma 2 +I ) 2 J (ma 2 +I ) ⎜ ⎟ ⎜ ⎟ (2.8) ω=⎜ ⎟ √ % % ⎜ √1 ⎟ 0 − √ 2 η2 ⎟ ⎜ − 2 J (mam2 +I ) η2 √12 J (mam2 +I ) η1 J ⎜ ⎟ ⎜ ⎟ ⎝ ⎠ √ 2 2 √ η 0 0 0 J

so, in particular, ω12 = −ω21 =

1 2

#

m η3 . J (ma 2 + I )

88


Let c : R → Q be a nonholonomic geodesic given by c(t) ˙ = v1 (t)X1 + v2 (t)X2 . From the structure equations we see immediately that ω12 (c(t)) ˙ = −ω21 (c(t)) ˙ =0 d d and the nonholonomic geodesic equations reduce to dt (v1 ) = dt (v2 ) = 0. The ˙ θ˙ ) = AX1 + BX2 . In particular, nonholonomic geodesics are solutions to (x, ˙ y, ˙ φ, √ √ 2Aa cos θ (t) 2Aa sin θ (t) x˙ = √ , y˙ = √ , ma 2 + I ma 2 + I (2.9) √ √ 2A 2B ˙ ˙ φ=√ , θ= √ . J ma 2 + I The trajectories are spinning in place (A = 0), rolling along a line (B = 0), or circles (A, B = 0). 2.2 Equivalence problem of nonholonomic geometry Cartan’s method of equivalence starts by encoding a geometric structure in terms of a subbundle of the coframe bundle called a G-structure. We begin this section by describing the G-structure for nonholonomic geometry16 . We then give a brief outline of some of the main ideas behind the method of equivalence as it is applied in our example of nonholonomic geometry on an Engel manifold. Details about the method of equivalence can be found in Gardner [1989], Montgomery [2002], or Bryant [1994]. We then derive the local invariants associated with a nonholonomic structure on a four-dimensional manifold endowed with an Engel distribution. Initial G-structure for nonholonomic geometry A coframe η(x) at x ∈ Qn is a basis for the cotangent space Tx∗ (Q). Alternatively, we can regard a coframe as a linear isomorphism η(x) : Tx (Q) → Rn where Rn is represented by column vectors. A coframe can then be multiplied by a matrix on the left in the usual way. The set of all coframes at x is denoted Fx∗ (Q) and has the projection mapping π : Fx∗ (Q) → x. The coframe bundle F ∗ (Q) is the union of the Fx∗ (Q) as x varies over Q.Acoframe on Q is a smooth (local) section η : Q → F ∗ (Q) and is represented by a column vector of 1-forms (η1 , . . . , ηn )tr , where “tr’’ indicates transpose. F ∗ (Q) is a right Gl(n)-bundle with action Rg η = g −1 η where g is a matrix in Gl(n). Let G be a matrix subgroup of Gl(n). A G-structure is a G-subbundle of F ∗ (Q). We now describe the G-structure encoding the nonholonomic geometry associated with a nonholonomic structure (Q, G, H). Given a nonholonomic structure (Q, G, H) we can choose an orthonormal coframe η = (ηi , ην )tr on U ⊂ Q so that the ην annihilate H and use this coframe to write down the nonholonomic geodesic equations as described above. On the other hand, given acoframe η¯ = (η¯ i , η¯ ν )tr on Q we can ¯ where H¯ is construct a nonholonomic structure (Q, G¯ = η¯ i ⊗ η¯ i + η¯ ν ⊗ η¯ ν , H) 16 This G-structure was first presented by Cartan in his 1928 address to the International

Congress of Mathematicians (Cartan [1928])


89

annihilated by the η¯ ν . How is η¯ related to η if it is to lead to the same nonholonomic geodesic equations as η? In order to preserve H we must have ην − η¯ ν = 0 (mod I ). In matrix notation, any modified coframe η¯ must be related to η by i i Ab η¯ η = , (2.10) 0 a η¯ ν ην where A ∈ Gl(r), a ∈ Gl(n − r), and b ∈ M(k, n − r). If we were studying the geometry of distributions, there would be no further restrictions. In order to preserve the metric restricted to H, we must further insist that A ∈ O(r). We would then have the starting point for the study of sub-Riemannian geometry (see Montgomery [2002], Hughen [1995], or Moseley [2001]). It is important to observe that in nonholonomic geometry we need the full metric and not just its restriction to H (as in sub-Riemannian geometry) to obtain the equations of motion. Cartan [1928] showed that in order to preserve the nonholonomic geodesic equations, we can only add covectors that are in the first derived ideal to the ηi . Since this fact is central to our analysis, we sketch the argument here (see Koiller, Rodrigues, and Pitanga [2001] for details). Suppose η¯ = gη with connection 1-form defined by d η¯ = −ω¯ ∧ η. ¯ For simplicity, assume that A = id; then ηj ≡ η¯ j (mod I). The geodesic equations are preserved if and only if ωij (T ) = ω¯ ij (T ) for all T ∈ H, in other words ωij ≡ ω¯ ij (mod I). Note also that η¯ ν ≡ 0(mod I). Subtracting the structure equations for dηi and d η¯ i , we get dηi − d η¯ i = −ωij ∧ ηj − ωiν ∧ ην + ω¯ ij ∧ η¯ j + ω¯ iν ∧ η¯ ν ≡ 0

(mod I).

Now η¯ i = ηi + biν ην so we also have dηi − d η¯ i = dηi − (dηi + dbiν ην + biν dην ) ≡ −biν dην

(mod I).

Therefore, biν dην ≡ 0 (mod I) or, equivalently, biν ην ∈ I (1) . This completes the argument. We further subdivide our indicial notation: let r +1≤φ ≤s

(= rank H1 ),

s + 1 ≤ ≤ n.

Adapted coframes A covector η = (ηi , ηφ , η )tr ) arranged so that 1. The ηφ and I, η i generate 2 2. ds |H = η ⊗ ηi , 3. The η generate the first derived ideal I (1) ,

is said to be adapted to the nonholonomic structure. In matrix notation, the most general change of coframes that preserves the nonholonomic geodesic equations is of the form η¯ = gη where

90


⎞ A 0 b g = ⎝ 0 a1 a2 ⎠ 0 0 a3 ⎛

(2.11)

with A ∈ O(k), b ∈ M(n − s, k), a1 ∈ Gl(s − k), a2 ∈ M(n − s, s − k), and a3 ∈ Gl(n − s). The set of all such block matrices form a matrix subgroup of Gl(n) which we shall denote G0 . The initial G-structure for nonholonomic geometry on (Q, ds 2 , H) is a subbundle B0 (Q) ⊂ F ∗ (Q) (or simply B0 if there is no risk of confusion) with structure group G0 defined above. All local sections of B0 (Q) lead to the same nonholonomic geodesic equations. In this way, the initial G-structure B0 (Q) completely characterizes the nonholonomic geometry. πQ

πN

Two G-structures, B(Q) → Q and B(N ) → N , are said to be equivalent if there is a diffeomorphism f : Q → N for which f1 (B(Q)) = B(N ) where f1 is the induced bundle map. (If we think of b ∈ B(Q) as a linear isomorphism b : TπQ (b) Q → Rn then f1 (b) = b ◦ (f∗ )−1 where f∗ is the differential of f .) Our original question as to whether there is a local diffeomorphism that carries nonholonomic geodesics to nonholonomic geodesics can be answered by determining whether the associated G-structures are locally equivalent. 2.3 A tutorial on the method of equivalence Necessary and sufficient conditions for the equivalence between G-structures are given in terms of differential invariants which are derived using the method of equivalence. In this section, we briefly describe some of the main ideas behind the method of equivalence as it is applied in our example. Details and other facets of the method together with many examples can be found in the excellent text by Robert Gardner (Gardner [1989]). One of the principal objects used in the method of equivalence is π the tautological 1-form. Let B(Q) → Q be a G-structure with structure group G whose Lie algebra is Lie(G). The tautological 1-form on B(Q) is an Rn -valued 1-form defined as follows. Let η : U ⊂ Q → B(Q) be a local section of B(Q) and consider the inverse trivialization U × G0 → B(Q) defined by (x, g) → g −1 η(x). Relative to this section, the tautological 1-form is defined by

(b) = g −1 (π ∗ η),

(2.12)

where b = g −1 η. From (2.12) one can verify that the tautological 1-form is semibasic (i.e., (v) = 0 for all v ∈ ker(π∗ )), has the reproducing property η¯ ∗ = η, ¯ where η¯ is any local section of B(Q), and is equivariant: Rg∗ = g −1 . The components of the tautological 1-form provide a partial coframing for B(Q) and form a basis for the semibasic forms on B(Q). The following proposition reduces the problem of finding an equivalence between G-structures to finding a smooth map that preserves the tautological 1-form. (See Gardner [1989] or Bryant [1994] for a proof.)


91

Proposition 2.1. Let B(Q) and B(N ) be two G-structures with corresponding tautological 1-forms Q and N , and let F : B(Q) → B(N ) be a smooth map. If G is connected and F ∗ ( N ) = Q , then there exists a local diffeomorphism f : Q → N for which F = f1 , i.e., the two G-structures are equivalent. To find the map F in this proposition we would like to apply Cartan’s technique of the graph (see Warner [1971], p. 75): if we could find an integral manifold ⊂ B(Q) × B(N ) of the 1-form θ = Q − N that projects diffeomorphically onto each factor, then would be the graph of a function h : Q → N for which h∗1 N = Q . By the above proposition the G-structures would then be equivalent. We generally cannot apply this idea directly because Q and N do not provide full coframes on B(Q) and B(N ) as is required in the technique of the graph. In the example of nonholonomic geometry on Engel manifolds, and indeed in many important examples (see Gardner [1989], Hughen [1995], Moseley [2001], Montgomery [2002], Ehlers [2002]), applying the method of equivalence leads to a new G-structure called an e-structure. An e-structure is a G-structure endowed with a canonical coframe. Differentiating both sides of (2.12) one can verify that d satisfies the structure equation d = −α ∧ + T , (2.13) where T is a semibasic 2-form on B(Q) and α is called a pseudoconnection: a Lie(G)valued 1-form on B(Q) that agrees with the Mauer–Cartan form on vertical vector fields. Here, Lie(G) is the Lie algebra of G. Summarizing, Pseudoconnection:

α = g −1 dg + semibasic Lie(G)-valued 1-form.

(2.14)

The components of the pseudoconnection together with the tautological 1-form do provide a full coframe on the G-structure, but unlike the tautological 1-form, the pseudoconnection is not canonically defined. Understanding how changes in the pseudoconnection affect the torsion is at the heart of the method of equivalence. For any G-structure, that part of the torsion that is left unchanged under all possible changes of pseudoconnection is known as the intrinsic torsion. The intrinsic torsion is the only first-order differential invariant of the G-structure (Gardner [1989]). As an example, the intrinsic torsion for the G-structure B of a general distribution (equation 2.10) is the dual curvature of the distribution (Cartan [1910], see also Montgomery [2002]). In the case of a rank two distribution on a four-dimensional manifold, the structure equations for the tautological 1-form are ⎛ ⎞ ⎞ ⎛ 1⎞ ⎛ 1⎞ ⎛

T

1 A11 A12 β13 β14 ⎜ 2 ⎟ ⎜ A21 A22 β23 β24 ⎟ ⎜ 2 ⎟ ⎜ T 2 ⎟ ⎟ ⎟ ⎜ ⎟ ⎜ ⎟ ⎜ d⎜ (2.15) ⎝ 3 ⎠ = − ⎝ 0 0 α33 α34 ⎠ ∧ ⎝ 3 ⎠ + ⎝ T 3 ⎠ ,

4 0 0 α34 α44

4 T4 where T I = J 3 the problem is open. For basic informations, see Fedorov and Kozlov [1995], pp. 147–149, on the 3D case and pp. 153–156 for the general n-dimensional case. For a detailed account of the algebraic integrability of “Chaplygin’s Chaplygin sphere’’; see Duistermaat [2000]. Schneider [2002] analyzed control theoretical aspects.

104


defined by D : z˙ = 0, x˙ = rω1 , y˙ = −rω2 . Both Lagrangian and constraints are preserved under the action of the Euclidean motions in the plane, together with the vertical translations. G = SE(2) × R acts on Q via (φ, u, v, w).(R, x, y, z) = (S(φ)R, eiφ (u + iv), z + w). The dynamics could be directly reduced to D/G (see, e.g., Zenkov and Bloch [2003]), but we will proceed in two stages. First, we Chaplygin-compress the dynamics from T Q to T SO(3) using the translation subgroup of SE(3), regarding the constraint distribution as an abelian connection on Q with base space S = SO(3) and fiber R3 ; the connection form is given by αmarble := (dx − rρ2 , dy + rρ1 , dz).

(3.18)

There is another S 1 action on Q, this time acting on the first factor only: eiφ (R, z) = (S(φ)R, z). This action preserves the Lagrangian but does not preserve the distribuiφ tion: D(S(φ)R,z) = e∗ D(R,z) . However, its infinitesimal action is given by the right vector field X3r ∈ D. Noether’s theorem applies, so pφ = 3 is a constant of motion. Therefore, Chaplygin’s marble equations can be reduced, on each level set 3 , to T (SO(3)/S 1 ) = T S 2 . In the case of Chaplygin’s rubber ball,20 rotations about the vertical axis are forbidden (since such rotations would cause energy dissipation). Here the constraints are defined by a subdistribution H ⊂ D with Cartan’s 2-3-5 growth numbers and, in fact, defining a connection on SE(2) × R → Q → S 2 with 1-form ˆ dx − rρ2 , dy + rρ1 , dz). αrubber := (ρ3 k,

(3.19)

The extrinsic viewpoint For clarity we present the classical, direct derivation of the equations of motion, following the “extrinsic viewpoint’’ advocated by the Russian Geometric Mechanics school (Borisov and Mamaev [2002a]). • For the rubber Chaplygin ball (and Veselova’s): in the space frame one has ˙ = τ , where τ = λkˆ is the torque exerted by the constraint force. The torque is vertical because (τ, ω) = 0 for all ω with third component equal to zero. Viewed in the body frame, L˙ + × L = λγ , (3.20) Together (1.6), one gets a closed system of ODEs in the space (L, γ ) ∈ R3 × R3 , provided the relation between and L is obtained. In Veselova’s example, = A−1 L. The multiplier can be eliminated by differentiating the constraint equation ( , γ ) = 0. After a simple computation, one gets 20 This problem was not studied by Chaplygin. For the physical justification, see Neimark and

Fufaev [1972] and Cendra, Ibort, de Léon, de Diego [2004]. As far as we know its integrability has not yet been established. Formally, Veselova’s system is the limit of Chaplygin’s rubber ball as r → 0.


λ=

(L, A−1 γ × A−1 L) . (γ , A−1 γ )

105

(3.21)

Besides the standard integrals of motion 2H = (A−1 L, L), (γ , γ ) = 1, (A−1 L, γ ) = 0, Veselov and Veselova [1988] showed that there is a quartic polynomial integral G = (L, L) − (L, γ )2

(3.22)

and an invariant measure21 µ = f (γ )dL1 ∧ dL2 ∧ dL3 ∧ dγ1 ∧ dγ2 ∧ dγ3 ,

f (γ ) = (A−1 γ , γ )−1/2 . (3.23)

• For Chaplygin’s marble: the angular momentum at the contact point in the space frame is constant. An engineer would argue that both gravity and friction produce no torque at that point; a mathematician would use the fact that the admissible vector fields Vi ∈ H given by right

V1 := −r∂/∂y + X1

,

right

V2 := r∂/∂x + X2

,

right

V3 := X3

(3.24)

preserve the Lagrangian, and would invoke NH-Noether’s theorem. Whichever explanation chosen, differentiating RL = = RL and Rγ = k, one gets Chaplygin’s equations L˙ = − × L, γ˙ = − × γ . (3.25) These two form a coupled system, since again is a linear function of L depending only on γ : ˜ − µr 2 (γ , )γ , L = Lγ ( ) = A + µr 2 γ × ( × γ ) = A

A˜ := A + µr 2 id. (3.26)

A simple way to get this map is to look at the total energy 2T = (ω, ) = ( , L) = (A , ) + µ(x˙ 2 + y˙ 2 ) = (A , ) + µr 2 (ω12 + ω22 ), (3.27) which can be also written as 2T = ( , L) = (A , ) + µr 2 ( , γ × ( × γ )) = ( , A + µr 2 γ × ( × γ ))). (3.28) The expression γ × (• × γ ) represents the projection in the plane perpendicular to γ , and we get (3.26). An ansatz for the inverse of the map (3.26) is (Duistermaat [2000]),

= (L, γ ) = (Lγ )−1 (L) = A˜ −1 L + α(L)A˜ −1 (γ ), (3.29) and one gets the interesting expression for α(L) (which will be used in equation (3.48) and Proposition 3.8): 21 The level sets of the four integrals are 2-tori, since there are no fixed points in the dynam-

ics. The existence of an invariant measure in the tori allows the explicit integration via Jacobi’s theorem. Veselov and Veselova [1988] found a “rather unexpected connection with Neumann’s problem.’’

106


α(L) = µr 2 The function

(γ , A˜ −1 L) . 1 − µr 2 (γ , A˜ −1 γ )

(3.30)

f (γ ) := [1 − µr 2 (γ , A˜ −1 γ )]−1/2

was found by Chaplygin to be the density of an invariant measure in

(3.31) R6 :

νR6 = f (γ )dγ1 dγ2 dγ3 dL1 dL2 dL3 .

(3.32)

This follows from Veselova’s theorem, as F (γ ) = 1 − µr 2 (γ , A˜ −1 γ ) is (up to a constant factor) the determinant of the linear map → L = L( ; γ ). For direct proofs of invariance of the measure, see Duistermaat [2000] or Fedorov and Kozlov [1995]. A system of ODE’s for the rubber ball can be derived in a similar fashion. For the angular momentum at the contact point, we get the same equation (3.20) from Veselova’s system, but the relation between and L is (3.26), the same as in Chaplygin’s marble. Differentiating ( , γ ) = 0 the multiplier can be eliminated. Hamiltonization of Veselova’s system The compressed Lagrangian is Lcomp =

1 (A(γ˙ × γ ), γ˙ × γ ), 2

(3.33)

since = γ˙ × γ ; the momentum map corresponding to the S 1 -action is J = 3 = (L, γ ). Thus (J.K) = 3 dρ3 = (A , γ )dρ3 , where dρ3 is the area form of S 2 . The compressed Legendre transform is γ˙ → a =

∂L∗ = γ × A(γ˙ × γ ). ∂ γ˙

The nonholonomic 2-form in T ∗ S 2 is

N H = da ∧ dγ + (A(γ˙ × γ ), γ )dρ3 .

(3.34)

Being a two-degrees of freedom system, a general result from Fedorov and Jovanovic [2003] (Theorem 3.5) guarantees that this system is Hamiltonizable. In order to verify that N H is conformally symplectic, it is simpler to use γ˙ as coordinates, that is, we pull back N H to T S 2 via Leg∗ . We get

N H = d(γ × A(γ˙ × γ ))) ∧ dγ + (γ , A(γ˙ × γ ))dρ3 . Proposition 3.5. Veselova’s system is conformally symplectic, d(f N H ) = 0, with conformal factor f = f (γ ) = (A−1 γ , γ )−1/2 . (3.35) As expected, it is the density of the Veselova invariant measure µ = f (γ )dLdγ obtained via Proposition 3.3. The orthonormal frame in S 2 diagonalizing (3.33) provides explicit coordinates for integration via the Hamilton–Jacobi method.


107

Chaplygin’s rubber ball The dynamics compress to T ∗ S 2 , and by the same general result in Fedorov and Jovanovic [2003], we know in advance that the system is Hamiltonizable. Choose a moving frame e1 , e2 in S 2 . The horizontal lift from γ˙ = v1 e1 + v2 e2 to Hor(γ˙ ) ∈ T (SE(3)) is easily done via (1.10): Hor(γ˙ ) = v2 (X1r − r∂/∂y) − v1 (X2r + r∂/∂x). Composing dαrubber = (ρ1 ∧ ρ2, −rρ3 ∧ ρ1 , rρ2 ∧ ρ3 , 0) with Hor, we get Krubber = ˆ 0, 0, 0), where dS is the S 2 area form. Thus for the term (J.K) we need only (dS k, the third component of the angular momentum, m3 = (M, γ ) = (A , γ ), where we insert (1.10) = γ˙ × γ = v2 e1 − v1 e2 . Therefore,

N H = T ∗ S 2 + (A(γ˙ × γ ), γ ) · dS.

(3.36)

Here γ˙ = v1 e1 + v2 e2 ∈ T S 2 corresponds to pγ = p1 θ1 + p2 θ2 via the Legendre map Legcomp of the compressed Lagrangian Lcomp =

1 1 A(v2 e1 − v1 e2 , v2 e1 − v1 e2 ) + µr 2 (v12 + v22 ). 2 2

(3.37)

Clearly, this system becomes Veselova for r = 0. Using Proposition 3.3 and Fedorov’s result for two degrees of system, we get Proposition 3.6. Proposition 3.6. The compressed rubber ball system is Hamiltonizable. The conformal factor is f = [det Legcomp ]−1/2 '

= (I1 I2 I3 )−1/2 (A−1 γ , γ ) + µr 2

(

γ22 + γ33 I2 I3

)

γ 2 + γ33 γ 2 + γ23 µ2 r 4 + + 1 + 1 I1 I3 I1 I2 I1 I2 I3

(3.38)

*−1/2

.

Proof. We checked using spherical coordinates and MathematicaTM .22 3.3 Chaplygin’s marble is not Hamiltonizable at the T ∗ SO(3) level The homogeneous sphere In a nutshell, the dynamics in the homogeneous case are embarrassingly simple. The angular velocity in space is constant, so the attitude matrix R evolves as a oneparameter group R = exp([ω]t), so and ω are constant. The vector γ (t) describes a circle in the sphere perpendicular to ω, and L(t) the curve given by L(t) = (I + µr 2 )ω − ω3 γ (t). Provided is not vertical, L and γ are never parallel. The invariant tori are always foliated by closed curves and the two frequencies coincide. From 22 We can provide the (short) notebook under request. It should be investigated if the rubber

ball problem is integrable. Does a (quartic) integral still exist?

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the constraint equations we see that the motion of the contact point in the plane is a straight line. Shooting pool with a perfect Chaplygin ball is very dull.23 Let us use these simple results as template for our operational system. In terms of the right coframe, we have

N H = d1 ρ1 + d2 ρ2 + d3 ρ3 + 1 ρ2 ρ3 + 2 ρ3 ρ1 + 3 ρ1 ρ2 − µr 2 (ω2 ρ3 ρ1 + ω1 ρ2 ρ3 ).

(3.39)

This formula holds in general. In the nonhomogeneous case one must write ω1 and ω2 in terms of and R ∈ SO(3): ω = R = R γ (R −1 ) which seems to be a quite involved expression, a haunting monster we will avoid, until a final confrontation in Proposition 3.8. In the homogeneous case, life is much easier: ω = R κ1 I R −1 m = I1 m, so the dependence of ω on R disappears. The Hamiltonian is given by * ' 2 1 21 + 22 H = + 3, 2 2 I + µr I where

µr 2 1 = 1 + m1 , I m1 ω1 = , I

µr 2 2 = 1 + I m2 ω2 = , I

To obtain the equations of motion we solve ⎛ ⎞ ⎛ ω1 0 0 0 1 ⎜ ω2 ⎟ ⎜ 0 0 0 0 ⎜ ⎟ ⎜ ⎜ ω3 ⎟ ⎜ 0 0 0 0 ⎜ ⎟=⎜ ⎜ ˙1 ⎟ ⎜ −1 0 0 0 ⎜ ⎟ ⎜ ⎝ ˙2 ⎠ ⎝ 0 −1 0 −3 0 0 −1 I ω2 ˙3

0 1 0 3 0 −I ω1

m2 ,

3 = m3 , ω3 =

m3 . I

⎞ ⎛ ⎞ 0 0 ⎟ ⎜0 ⎟ 0 ⎟ ⎜ ⎟ ⎟ ⎜0 ⎟ 1 ⎟ · ⎜ ⎟, ⎜ ⎟ −I ω2 ⎟ ⎟ ⎜ ω1 ⎟ ⎠ ⎝ ω2 ⎠ −I ω1 0 ω3

(3.40)

where we have used H1 = 1 /(I + µr 2 ) = m1 /I = ω1 , and similarly, H2 = ω2 , H2 = ω2 . This gives, as expected ˙1 = (I ω3 )H2 − I ω2 H3 = 0,

˙2 = · · · = 0,

˙3 = · · · = 0. right

Thus ωi = mi /I = const, i = 1, 2, 3, and the vector field is simply X = ω1 X1

+

23 We found the following relevant information in www.ot.com/skew/five/myths. html (Top

Ten Myths in Pool or the Laws of Physics Do Apply): “4. If the cue is kept level, contacting the cueball purely left or right of its center will make it curve as it rolls. (No! The rolling cue ball can have two completely independent components to its angular momentum. Basically, this means that it can rotate in the manner of a top while rolling slowly forward along a straight line. In general, spin on a cue ball is of two types; follow/draw is the spin like tires on a car, while English is the spin like a child’s toy ‘top.’ Separately, neither one will make a ball curve! If they are combined—e.g., strike low-left giving left English and draw—then the spin is called masse (“mass-ay’’), and the ball will curve as it travels.)’’

Nonholonomic systems via moving frames right

109

right

ω2 X2 + ω3 X3 (no components in the fiber directions ∂/∂mi ). We now use Theorem 3.4. Using m as coordinates, the nonholonomic 2-form is given by µr 2

N H = 1 + (dm1 ρ1 + dm2 ρ2 ) I + dm3 ρ3 + (m1 ρ2 ρ3 + m2 ρ3 ρ1 + m3 ρ1 ρ2 ) 2

so that d N H = − µrI (dm1 ρ2 ρ3 + dm2 ρ3 ρ1 ). It is easy to see that the equation d N H = N H ∧ α has no solution. Indeed, suppose α = A1 dm1 + A2 dm2 + A3 dm3 + B1 ρ1 + B2 ρ2 + B3 ρ3 . Taking the exterior product, and looking at terms like dm1 dm2 ρ2 we see that all the A’s must be zero. Examining the coefficient of ρ1 ρ2 ρ3 we get B1 m1 + B2 m2 + B3 m3 ≡ 0 so all the B’s are also zero. Hence the homogeneous Chaplygin sphere, as simple at it can be, has no conformal symplectic structure! In fact, it does not have an affine symplectic structure either. A short calculation shows that µr 2 (−dm1 m2 ρ3 + dm1 ρ2 m3 − dm2 m3 ρ1 + dm2 ρ3 m1 ) = 0. I2 By continuity, for sufficiently close but different inertia coefficients the inequalities persist. We have also done the calculation for the nonhomogeneous case and things only get worse. But, it still remains a possibility: is the reduced system to T ∗ S 2 Hamiltonizable? The impatient reader can go directly to Theorem 3.8. iX d N H =

3.4 Chaplygin’s marble: Reduction to T ∗ S 2 Using (1.8), L = a × γ + 3 γ , Chaplygin’s marble equations in (L, γ )-space directly reduce to T ∗ S 2 : γ˙ = γ × ,

a˙ = −2H γ + (γ , ) · (a × γ + 3 γ )

with

= (a, γ ; 3 ) = A˜ −1 L + µr 2

(3.41)

(γ , A˜ −1 L) A˜ −1 (γ ). 2 −1 ˜ 1 − µr (γ , A γ )

S 1 reduction of the homogeneous sphere to T ∗ S 2 The homogeneous Chaplygin sphere when reduced to T ∗ S 2 produces a more interesting system. Equations (3.41) become γ˙ =

1 a, I + µr 2

a˙ = ω3 a × γ −

1 |a|2 γ . I + µr 2

(3.42)

One observes that (a, γ ) = 0 and that |a|2 is conserved. So at each level set, we get an isotropic 3D oscillator with a Lorentz force.24 24 Alan Weinstein commented on more than one occasion that “unreduction’’ sometimes is

even nicer than reduction: unreducing a nontrivial system may lead to a trivial one. Alan credits this to Guillemin and Sternberg; one reference could be Guillemin and Sternberg [1980].

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Dimension count argument In hindsight, we can give two simple arguments why the Chaplygin marble could not be Hamiltonizable at the T ∗ SO(3) level. First, if (T ∗ SO(3), N H , H ) were Hamiltonizable, the system would be Liouville integrable by “mere’’symmetries, due to the existence of three independent first integrals H, 3 , 21 + 22 , 23 . But it is known that integrability of Chaplygin’s marble stems not from symmetries, but from a special choice of separating coordinates (Duistermaat [2000]), namely, elliptic coordinates on the sphere. Second, Stanchenko [1985] verified that Chaplygin’s density function F (3.31) of the system in R6 also gives an invariant measure on T ∗ SO(3) (see also Duistermaat [2000], Section 7), F = [1 − µr 2 (γ , A˜ −1 γ )]−1/2 . (3.43) Were the compressed system Hamiltonizable in T ∗ SO(3), the conformal factor (time 1 reparametrization) would be F (γ ) m−1 , with m = 3; see (3.13). But the correct time reparametrization holds with m = 2 instead of m = 3. This strongly suggests that Hamiltonization should be attempted after reduction of the internal S 1 symmetry. νT ∗ SO(3) = F (γ )dλ1 dλ2 dλ3 dL1 dL2 dL3 ,

Phase locking The fact that Chaplygin’s sphere is integrable implies an interesting phase locking property. For simplicity, consider a resonant torus and a periodic solution, γ (T ) = γ (0), L(T ) = L(0). We may assume that R(0) = identity, so R(T ) preserves both k and . If we assume = ±k, then R(T ) must also be the identity (there is only one orthogonal matrix with two different eigenvectors with equal eigenvalues 1). Since the rotational conditions are reproduced after time T , there is a “planar geometric phase’’ (meaning a translation), z = ( x, y). From Duistermaat [2000], Section 11, one knows this direction. Proposition 3.7. On average,

z moves in the direction of × k.

In the normal direction k ×(×k) there is a “swaying motion,’’ with zero average, see Duistermaat [2000], (11.71), and Remark 11.11. This result depends on the explicit solution in terms of elliptic coordinates, but the zero average can be proved in a more elementary way, see Duistermaat, Section 8.2. In the direction × k one has d (z(t), × k) = r(ω × k, × k) = r(ω, − 3 k) = r(2T − 3 ω3 ) > 0. dt Duistermaat [2000] shows (in Section 9.2) that by a suitable change of coordinates, one may assume that 3 = 0, so in this equivalent problem, the velocity in this direction is simply 2rT . Chaplygin’s marble via the almost Hamiltonian structure After this detour, we hope the reader will appreciate a concise way of describing this system. The clockwise map is

Nonholonomic systems via moving frames T (SO(3) × R2 )

−→ Leg

T ∗ (SO(3) × R2 ) ( , x, ˙ y) ˙ → (M = A , Px = µx, ˙ Py = µy) ˙

↑ h | T SO(3)

111

↑ h | ←−

(Legφ )−1

T ∗ SO(3)

←

L,

(3.44) where (x, ˙ y) ˙ = rω × k, and (Px , Py ) = µrω × k. We now compute the “gyroscopic’’ 2-form (J.K) = r(−Px dρ2 + Py dρ1 ) = µr(−xdρ ˙ 2 + ydρ ˙ 1 ) = −µr 2 (ω2 dρ2 + ω1 dρ1 ). (3.45) To obtain ω1 and ω2 as functions in T ∗ SO(3), we use the Legendre transformation: ω = R = RA−1 M, so (J.K) is a combination of the basic forms ρ3 ∧ ρ1 , ρ2 ∧ ρ3 (coefficients linear in M and functions of R). S 1 invariance We claim that N H is S 1 -invariant (S 1 acting only in the first factor of Q = SO(3) × R3 ). For the canonical term this is a standard symplectic fact. The (J.K) term is invariant as well: (3.45), written in terms of the left-invariant forms, depends only on the Poisson vector γ : (J.K) = µr 2 (γ × ( (L, γ ) × γ ), dλ) .

(3.46) right

In fact, the S 1 action generated by the right-invariant vector field X3 maintains the projection γ fixed. We know (general nonsense) that the right-invariant vector fields ˙ = λi (Rφ R[ ]) = preserve the left-invariant forms: Rφ∗ λi = λi . (Proof: (Rφ∗ λi )(R) 1

i .) Since under the left S action (actually under the left action of SO(3) on SO(3)) the value of remains unchanged, the (J.K) term is preserved. The twisted action generator and S 1 reduction MW reduction method works fine, although X3r is the Hamiltonian vector field of J = 3 , relative to the canonical symplectic form, but not relative to N H . We just change to the twisted S 1 -action generator X˜ 3 , defined by iX˜ 3 N H = −d3 . A simple computation gives X˜ 3 = Xr − m2 ∂ + m1 ∂ , where m1 = 1 − µr 2 ω1 , 3

∂1

∂2

m2 = 2 − µr 2 ω2 . The reduced manifold is the quotient of a level 3 in T ∗ SO(3), ˜ A concrete realization is achieved using (1.11). Taking identifying the flow lines φ. ∗ the pullback via i , the reduced form is then

red = can + 3 areaS 2 − µr 2 (ω1 dθ2 − ω2 dθ1 ), T ∗S2

(3.47)

where we recall the parametrizations p1 θ1 + p2 θ2 ∈ T ∗ S 2 , R(γ ) = rows(e1 , e2 , γ ).

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In (3.47) we must write ω1 , ω2 explicitly in terms of p1 , p2 , 3 . To write this explicitly, there is no other option than to confront the monster (which actually is not that terrible): from = R −1 ω = ω1 e1 + ω2 e2 + ω3 γ and (3.26), we get ω = R(γ ) γ [R(γ )]† ,

= (p2 , −p1 , 3 ),

(3.48)

where γ is explicitly given by (3.30). Theorem 3.8. iX d(f red ) = 0, f (γ ) = [1 − µr 2 (γ , A˜ −1 γ )]−1/2 . Proof. We used spherical coordinates (fâute de mieux) and a MathematicaTM notebook. It misses being conformally symplectic by very little (even in the homogeneous case).25 Our calculation shows that Chaplygin’s sphere is not affine symplectic even at the T ∗ S 2 level, so Chaplygin’s sphere integrability is due to a specific nonholonomic phenomenon. This observation is in accordance with the opening statement in Duistermaat [2000]: “Although the system is integrable in every sense of the word, it neither arises as a Hamiltonian system, nor is the integrability an immediate consequence of the symmetries.’’

4 Recent developments and final comments NH systems have a reputation of having peculiar (even rebellious) dynamic behavior (Arnold, Kozlov, and Neishtadt [1988]). In spite of good progress, the general theory for NH systems is way behind the theory of Hamiltonian systems. For instance, although the groundwork for a Hamilton–Jacobi theory for NH systems has been set up in Weber [1986], not much has been achieved since. We have no intention (or competence) to make a survey of recent developments in NH systems, especially regarding reduction of symmetries; nevertheless it may be worth registering the intense activity going on. Recent books of interest are Cushman and Bates [1997], Cortés [2002], Oliva [2002], Bloch [2003] and a treatise in the mechanical engineering tradition is Papastavridis [2002].26 Reports on Mathematical Physics has been publishing NH papers regularly, and Regular and Chaotic Dynamics devoted large parts of vols. 1/2 (2002) to NH systems. For older eastern European literature, see P. M. M. USSR, J. Appl. Math. Mechanics, which has strongly influenced Chinese mechanics as well. For a historical account of NH systems, from a somewhat “antireductionist’’ perspective, see Borisov and Mamaev [2002a]. 25 Borisov and Mamaev [2002] showed by a subtle numerical evidence that, in the original time,

Chaplygin’s marble is not Hamiltonizable at any level of reduction. The question whether Chaplygin’s marble is Hamiltonizable in the new time dt/dτ = f (γ ) was addressed in Borisov and Mamaev [2001]. They provide a bracket structure in terms of the coordinates ˜ γ ), with L˜ = L/f (γ ). Using a computer algebra program we (L, γ ) or the coordinates (L, checked that the second brackets satisfy the Jacobi identity. However, we could not recover Chaplygin’s equations for the L coordinates, even in the homogenous case. 26 Reviewed in Koiller [2003].


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4.1 Invariant measures and integrability Kupka and Oliva [2001] and Kobayashi and Oliva [2003] find conditions ensuring a special, but very interesting situation, where the Riemann measure in T Q induced by the metric in Q is an invariant measure for the NH system. Invariant measures for systems with distributional symmetries were characterized in Zenkov and Bloch [2003]. Curiously, although a number of interesting NH systems have been solved using Abelian functions, a precise definition for integrability of a NH system is still lacking (Bates and Cushman [1999]). These examples suggest that the presence of an invariant measure must be imposed as a necessary (although not sufficient) condition for integrability (whatever it may be), see Kozlov [2002]. Most of them have enough integrals of motion that the dynamics occur on invariant two-dimensional tori. Due to the invariant measure, the flow becomes linear in these tori after a time rescaling. This follows from Jacobi’s multiplier method and Kolmogorov’s theorem (Arnold [1989]). Time reparametrization indicates the possibility of an affine symplectic structure. We believe that characterizing NH systems possessing an affine symplectic structure (if needed, after some reduction stage) could be an interesting project. As a first step, one may examine the existing literature to see which examples fit. We list a few papers for that purpose: Veselov and Veselova [1988], Veselov and Veselova [1986], Fedorov [1989], Cushman, Hermans, and Kemppainen [1995], Zenkov [1995], Zenkov and Bloch [2000], Dragovic, Gajic´ , and Jovanovic [1998], Jovanovic [2003], Fedorov and Jovanovic [2003]. One can hope that the manifestly geometric character of (1.14) can be instrumental to understand when, where and why Hamiltonization is possible. Moreover, a prior geometric understanding of the invariant volume form conditions is a more general question. It would be also interesting to tie the “Hamiltonizable’’ question with the invariants from the Cartan equivalence viewpoint, see below. 4.2 Nonholonomic reduction ´ The difficulties in reduction for general NH systems are explained in Sniatycki [2002]. There are four current theories of reduction of symmety for nonholonomic systems27 : (i) projection methods; see Marle [1995], Dazord [1994]; (ii) the distributional Hamiltonian approach, initiated by Bocharov and Vinogradov ´ [1977] and developed in Bates and Sniatycki [1993], Cushman, Kemppainen, ´ ´ ´ Sniatycki, and Bates [1995], Sniatycki [1998], and Cushman and Sniatycki [2002]. (iii) bracket methods, initiated by Mashke and van der Schaft [1994], and developed by Koon and Marsden [1998] and Sn´ iatycki [2001]; (iv) Lagrangian reduction; see Cendra, Marsden, and Ratiu [2001]. A few other references in this rapidly developing theme, besides those already mentioned are Bates [2002], Koon and Marsden [1997], Cantrijn, de Léon, Marrero, and de Diego [1998], Cortés and de Léon [1999], Marle [1998], Marle [2003]. 27 We thank one of the referees for this information.

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Almost Poisson, almost Dirac approaches Mashke and van der Schaft [1994] were the first to describe a NH system using an almost-Poisson structure,28 x˙i = {xi , H }MS . This bracket, defined on the manifold P = Leg(H) ⊂ T ∗ Q, where Leg : T Q → T ∗ Q is the Legendre transformation, in general does not satisfy the Jacobi identity. They proved that the Jacobi identity holds if and only if the constraints are integrable. In Koiller, Rios, and Ehlers [2002] we gave a moving frames based derivation of the bracket structure. For some recent work on the MS-bracket and also Dirac estructures (the latter introduced in Courant [1990]), see Cantrijn, de Léon, de Diego [1999], Koon and Marsden [1998], Ibort, de Léon, Marrero, and de Diego [1999], Clemente-Gallardo, Maschke, and van der Schaft [2001]. In spite of these advances, a complete understanding of the NH bracket geometry is still in order.29 4.3 G-Chaplygin systems via affine connections Trajectories of the compressed system can be described as geodesics of an affine connection ∇ N H in S (Vershik and Fadeev [1981], Koiller [1992]). For background in this approach, see Lewis [1998] and references therein. Consider the parallel transport operator along closed curves; if the holonomy group is always conjugate to a subgroup of S0(m), then the connection is metrizable. This means that there is a metric such that ∇ N H is precisely the Levi-Civita connection of this metric. More generally, one may want to know when the geodesics of ∇ N H are, up to time reparametrization, the geodesics of a Riemannian metric. This is a traditional area in differential geometry, whose roots go back to the 19th century, and goes under the name of projectively equivalent connections (Cartan [1937], Eisenhart [1925], Kobayashi and Nomizu [1963], Sharpe [1997]). Grossman [2000] studies integrability of geodesics equations via the equivalence method. Our problem, then, is to find conditions for the NH connection to be projectively equivalent to a Riemannian connection. It would be also interesting to tie the Hamiltonization question with the canonical system and invariants of the Cartan equivalence method. When an internal symmetry group is present, it would be desirable to construct a projected connection in S for each set of conserved momenta, and address these issues in the reduced level. Acknowledgments Our thanks to Hans Duistermaat for information on Chaplygin’s sphere and the referees for very good criticism and suggestions. This is also a special occasion to thank our mathematical family: Alan, of course; mathematical brothers and sisters from all continents (especially Yilmaz Akyildyz and Henrique Bursztyn) and cousins (especially Tudor Ratiu and 28 Physicists are never shy to use the word “super’’ in their endeavors; on the other hand we,

mathematicians, prefer to use low-key terminology, like “almost-quasi-twisted-(freakaz-)‘oid’s’’; this certainly does not help our image problem with applied people, see Papastavridis [2002] and Koiller [2003]. 29 Observations by J. Marsden (joint work with H. Yoshimura), and by C. Marle in their Alanfest talks are important steps in this direction.


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Debra Lewis), “uncle’’ Jerry Marsden, and, last but not least, “grandfather’’ Chern (with his gentle voice, commanding us to keep interested in Math, up to his age). We shall toast in many more Alanfests: Madadayo!

References Abraham, R., Marsden, J. [1994], Foundations of Mechanics, 2nd revised ed., Perseus Publishing, Boulder, CO. Arnold, V. I. [1989], Mathematical Methods of Classical Mechanics, 2nd ed., Graduate Texts in Mathematics, Vol. 60, Springer-Verlag, New York; 1st ed., 1978. Arnold, V. I., Kozlov, V. V., Neishtadt, A. I. [1988], Mathematical aspects of classical and celestial mechanics, in Arnold, V. I., ed., Dynamical Systems III, SpringerVerlag, New York. Bates, L. [2002], Problems and progress in nonholonomic reduction, Rep. Math. Phys., 49:2–3, 143–149. Bates, L., Cushman, R. [1999], What is a completely integrable nonholonomic dynamical system?, Rep. Math. Phys., 44:1–2, 29–35. ´ Bates, L., Sniatycki, J. [1993], Nonholonomic reduction, Rep. Math. Phys., 32:1, 99–115. Blackall, C. J. [1941], On volume integral invariants of non-holonomic dynamical systems, Amer. J. Math., 63:1, 155–168. Bloch, A. M. [2003], Nonholonomic Mechanics and Control, Springer-Verlag, New York. Bloch, A. M., Krishnaprasad, P. S., Marsden, J. E., Murray, R. M. [1996], Nonholonomic mechanical systems with symmetry, Arch. Rational Mech. Anal., 136, 21–99. Bocharov, A. V., Vinogradov, A. M. [1977], The Hamiltonian form of mechanics with friction, nonholonomic mechanics, invariant mechanics, the theory of refraction and impact, Appendix II in Kuperschmidt, B. A. and Vinogradov, A. M., “The structure of Hamiltonian mechanics,’’ Russian Math. Surveys, 42:2, 177–243. Borisov, A. V., Mamaev, I. S. [2001], Chaplygin’s ball rolling problem is Hamiltonian, Math. Notes (Mat. Z.), 70:5, 793–795. Borisov, A. V., Mamaev, I. S. [2002], Obstacle to the reduction of nonholonomic systems to the Hamiltonian form, Dokl. Phys. USSR, 47:12, 892–894. Borisov, A. V., Mamaev, I. S. [2002a], On the history of the development of the nonholonomic dynamics, Regular Chaotic Dynam., 7:1, 43–47. Borisov, A. V., Mamaev, I. S. [2002a], The rolling body motion of a rigid body on a plane and a sphere: Hierarchy of dynamics, Regular Chaotic Dynam., 7:2, 177–200. Borisov A. V., Mamaev I. S., Kilin A. A. [2002], The rolling motion of a ball on a surface: New integrals and hierarchy of dynamics, Regular Chaotic Dynam., 7:2, 201–218. Bryant, R. [1994], Lectures on the Geometry of Differential Equations, Fall 1994 André Aisenstadt Lectures, Centre de Recherche Mathématique, Montreal, in preparation; unpublished lecture notes available at http://www.cimat.mx/gil.

116


Cantrijn, F., de Léon, M., Marrero, J. C., de Diego, D. [1998], Reduction of nonholonomic mechanical systems with symmetries, Rep. Math. Phys., 42:1–2, 25–45. Cantrijn, F., de Léon, M., de Diego, D. [1999], On almost-Poisson structures in nonholonomic mechanics, Nonlinearity, 12, 721–737. Cantrijn, F., Cortés, J., de Léon, M., de Diego, D. [2002], On the geometry of generalized Chaplygin systems, Math. Proc. Cambridge Philos. Soc., 132, 323–351. Cartan, É. [1910], Le système de Pfaff à cinq variables et les équations aux dérivées partielles du second ordre, Ann. Sci. École Norm., 27:3, 109–192. Cartan, É. [1926], La théorie des groupes finis et continus et la géométrie différentielle, traitées par la méthode du repère mobile: Leçons professées à la Sorbonne (rédigées par Jean Leray), Gauthier-Villars, Paris, 1951. Cartan, É. [1928], Sur la represéntation géométrique des systèmes matériels non holonomes, Proc. Internat. Congr. Math. Bologna, 4, 253–261. Cartan, É [1937], Leçons sur la théorie des espaces a connexion projective, GauthierVillars, Paris. Cartan, É. [2001], Riemannian Geometry in an Orthogonal Frame: From Lectures Delivered by Élie Cartan at the Sorbonne in 1926–27, World Scientific, River Edge, NJ, 2001 (translated from the 1960 Russian edition by Vladislav V. Goldberg; foreword by S. S. Chern; preface to the Russian edition by S. P. Finikov). Cendra, H., Lacomba, E. A., Reartes, W. [2001], The Lagrange-d’Alembert-Poincaré equations for the symmetric rolling sphere, in Proceedings of the 6th Dr. Antonio A. R. Monteiro Congress of Mathematics (Bahía Blanca, 2001), 19–32, Departamento de Matemática, Instituto de Matemática, Universidad Nacional del Sur, Bahía Blanca, Argentina; MR1919465 (2003g:70021). Cendra, H., Marsden, J. E., Ratiu, T. S. [2001], Geometric mechanics, Lagrangian reduction and nonholonomic systems, in Enguist, B., and Schmid, W., eds., Mathematics Unlimited: 2001 and Beyond , Springer-Verlag, New York, 221–273. Cendra, H., Ibort, A., de Léon, M., de Diego, D. [2004] A generalization of Chetaev’s principle for a class of higher order non-holonomic constraints, J. Math. Phys., submitted. Chaplygin, S. A. [1911], On the theory of the motion of nonholonomic systems: Theorem on the reducing factor, Mat. Sb., 28, 303–314. Chaplygin, S. A. [1981], Selected Works on Mechanics and Mathematics, Nauka, Moscow. Chaplygin, S. A. [2002], On a ball’s rolling on a horizontal plane, Regular Chaotic Dynam., 7:2, 131–148; original paper in Math. Sb., 24 (1903), 139–168. Bryant, R. L., Chern, S. S., Gardner, R. B., Goldschmidt, H. L., and Griffiths, P. A. [1991], Exterior Differential Systems, Mathematical Sciences Research Institute Publications, Vol. 18, Springer-Verlag, New York. Clemente-Gallardo, J., Mashke, B., van der Schaft, A. J. [2001], Kinematical constraints and algebroids, Rep. Math. Phys., 47:3, 413–429. Cortés, J. [2002], Geometric, Control and Numerical Aspects of Nonholonomic Systems, Springer-Verlag, New York. Cortés, J., de Léon, M. [1999], Reduction and reconstruction of the dynamics of nonholonomic systems, J. Phys. A Math. Gen., 32, 8615–8645.


117

Cortés, J., de Léon, M., de Diego, D., Martínez, S. [2003], Geometric description of vakonomic and nonholonomic dynamics: Comparison of solutions, SIAM J. Control Optim., 41:5, 1389–1412. Courant, T. J. [1990], Dirac manifolds, Trans. Amer. Math. Soc., 319:2, 631–661. Cushman, R., Hermans, J., Kemppainen, D. [1995], The rolling disk, in Nonlinear Dynamical Systems and Chaos, Progress in Nonlinear Differential Equations and Their Applications, Vol. 19, 21–60, Birkhäuser, Basel. ´ Cushman, R., Kemppainen, D., Sniatycki, J., Bates, L. [1995], Geometry of nonholonomic constraints, Rep. Math. Phys., 36:2–3, 275–286. Cushman, R., Bates, L. [1997], Global Aspects of Classical Integrable Systems, Birkhäuser, Basel, 1997. ´ Cushman, R., Sniatycki, J. [2002], Nonholonomic reduction for free and proper actions, Regular Chaotic Dynam., 7, 61–72. Dazord, P. [1994], Mécanique hamiltonienne en présence de contraintes, Illinois J. Math., 38, 148–175. Dragovic´ , V., Gajic´ , B., Jovanovic´ , B. [1998], Generalizations of classical integrable nonholonomic rigid body systems, J. Phys. A, 31:49, 9861–9869. Duistermaat, J. J. [2000], Chaplygin’s sphere, in Cushman, R., Duistermaat, J. J., ´ and Sniatycki, J., Chaplygin and the Geometry of Nonholonomically Constrained Systems, in preparation; arXiv.org/abs/math.DS/0409019. Eisenhart, L. P. [1925], Riemannian Geometry, Princeton University Press, Princeton, NJ; 5th printing, 1964. Ehlers, K. [2002], The geometry of nonholonomic three-manifolds, in Proceedings of the 4th International Conference on Dynamical Systems and Differential Equations, University of North Carolina at Wilmington, Wilmington, NC. Fedorov, Yu. N. [1989], Two integrable nonholonomic systems in classical dynamics, Vestnik Moskov. Univ. Ser. I Mat. Mekh., 4, 38–41 (in Russian). Fedorov, Yu. N., Kozlov, V. V. [1995], Various aspects of n-dimensional rigid body dynamics, in Kozlov, V. V., ed., Dynamical Systems in Classical Mechanics, AMS Translations (Series 2), Vol. 168, AMS, Providence, RI. Fedorov, Yu. N., Jovanovic, B. [2003], Nonholonomic LR systems as generalized Chaplygin systems with an invariant measure and geodesic flows on homogeneous spaces, J. Nonlinear Sci., to appear; arXiv: math-ph/0307016. Flanders, H. [1963], Differential Forms with Applications to the Physical Sciences, Academic Press, New York. Gardner, R. [1989], The Method of Equivalence and its Applications, SIAM, Philadelphia. Grossman, D. A. [2000], Torsion-free path geometries and integrable second order ODE systems, Selecta Math. (N.S.), 6, 399–442. Guillemin, V., Sternberg, S. [1980], The moment map and collective motion, Ann. Phys., 1278, 220–253. Hamel, G. [1949], Theoretische Mechanik: Eine einheitliche Einführung in die gesamte Mechanik, revised ed., Grundlehren der Mathematischen Wissenschaften, Vol. 57, Springer-Verlag, Berlin, New York, 1978.

118


Haller, S., Rybicki, T. [1999], On the group of diffeomorphisms preserving a locally conformal symplectic structure, Ann. Global Anal. Geom., 17, 475–502. Haller, S., Rybicki, T. [2001], Symplectic reduction for locally conformal symplectic manifolds, J. Geom. Phys., 37, 262–271. Hertz, H. [1899], The Principles of Mechanics Presented in a New Form by Heinrich Hertz, with an Introduction by H. von Helmholtz, Macmillan, London, New York. Hicks, N. J. [1965], Notes on Differential Geometry, Van Nostrand, New York. Hughen, K. [1995], The Geometry of Sub-Riemannian Three-Manifolds, Ph.D. thesis, Duke University, Durham, NC. Ibort,A., de Léon, M., Marrero, J. C., de Diego, D. [1999], Dirac brackets in constraind dynamics, Fortschr. Phys., 47:5, 459–492. Iliyev, Il. [1985], On the conditions for the existence of the reducing Chaplygin factor, P. M. M. USSR, 49:2, 295–301. Jovanovic, B. [2003], Some multidimensional integrable cases of nonholonomic rigid body dynamics, Regular Chaotic Dynam., 8:1, 125–132. Kazarian, M. R., Montgomery, R., Shapiro, B. [1997], Characteristic classes for the degenerations of two-plane fields in four dimensions, Pacific J. Math., 179:2, 355– 370. Kobayashi, S., Nomizu, K. [1963], Foundations of Differential Geometry, Vol. 1, Wiley, New York, London. Kobayashi, M. H., Oliva, W. M. [2003], A note on the conservation of energy and volume in the setting of nonholonomic mechanical systems, Qual. Theory Dynam. Systems, 5 (2004), 255–283. Koiller, J. [1992], Reduction of some classical non-holonomic systems with symmetry, Arch. Rational Mech. Anal., 118, 113–148. Koiller, J., Rodrigues, P. R., Pitanga, P. [2001], Nonholonomic connections following Élie Cartan, An. Acad. Brasileira Ciencias, 73:2, 165–190. Koiller, J., Rios, P. M. [2001], Nonholonomic systems with symmetry allowing a conformally symplectic reduction, in Delgado, J., Lacomba, E. A., and Pérez-Chavela, E., eds., Proceedings of the 4th International Symposium on Hamiltonian Systems and Celestial Mechanics (Mexico 2001), Kluwer, Dordrecht, the Netherlands, to appear; arXiv: math-ph/0203013. Koiller, J., Rios, P. M., Ehlers, K. [2002], Moving frames for cotangent bundles, Rep. Math. Phys., 49:2–3, 225–238. Koiller, J. [2003], Analytical Mechanics, Bull. Amer. Math. Soc. (N.S.), 40:3, 405– 419. Koon, W. S., Marsden, J. E. [1997], The Hamiltonian and Lagrangian approaches to the dynamics of nonholonomic systems, Rep. Math. Phys., 40, 21–62. Koon, W. S., Marsden, J. E. [1998], Poisson reduction for nonholonomic mechanical systems with symmetry, Rep. Math. Phys., 42, 101–134. Kozlov, V. V. [2002], On the integration theory of equations of nonholonomic mechanics, Regular Chaotic Dynam., 7:2, 161–176. Kummer, M. [1981], On the construction of the reduced phase space of a Hamiltonian system with symmetry, Indiana Univ. Math. J., 30, 281–291.


119

Kupka, I., Oliva, W. M. [2001], The Non-Holonomic Mechanics, J. Differential Equations, 169, 169–189. Levi, M. [1996], Composition of rotations and parallel transport, Nonlinearity, 9, 413–419. Lewis, A. D. [1998], Affine connections and distributions with applications to nonholonomic mechanics, Rep. Math. Phys., 42:1–2, 135–164. Marle, C. M. [1995], Reduction of constrained mechanical systems and stability of relative equilibria, Comm. Math. Phys., 174, 295–318. Marle, C. M. [1998], Various approaches to conservative and nonconservative nonholonomic systems, Rep. Math. Phys., 42:1–2, 211–229. Marle, C. M. [2003], On symmetries and constants of motion in Hamiltonian systems with nonholonomic constraints, Banach Center Publ., 59, 223–242. Marsden, J. E., Weinstein, A. [2001], Reduction of symplectic manifolds with symmetry, Rep. Math. Phys., 5, 121–130. Marsden, J. E., Weinstein, A. [2001], Some comments on the history, theory, and applications of symplectic reduction, in Landsman, N. P., and Pflaum, M., eds., Quantization of Singular Symplectic Quotients, Birkhäuser, Boston, 2001. Montgomery, R. [1991], How much does the rigid body rotate? A Berry’s phase from the 18th century, Amer. J. Phys., 59:5, 394–398. Montgomery, R. [2002], A Tour of Sub-Riemannian Geometries, Their Geodesics, and Applications, Mathematical Surveys and Monographs, Vol. 91, AMS, Providence, RI. Moseley, K. [2001], The Geometry of Sub-Riemannian Engel Manifolds, Ph.D. thesis, Duke University, Durham, NC, 2001. Neimark, J. I., Fufaev, N.A. [1972], Dynamics of Nonholonomic Systems, Translations of Mathematical Monographs, Vol. 33, AMS, Providence, RI. Oliva, W. M. [2002], Geometric Mechanics, Lecture Notes in Mathematics 1798, Springer-Verlag, New York. Papastavridis, J. G. [2002], Analytical Mechanics: A Comprehensive Treatise on the Dynamics of Constrained Systems: For Engineers, Physicists and Mathematicians, Oxford University Press, Oxford, UK (reviewed in Koiller [2003]). Pars, L. A. [1965], A Treatise on Analytical Dynamics, Wiley, New York. Poincaré, H. [1901], Sur une forme nouvelle des équations de la mécanique, C. R. Acad. Sci. Paris, 132, 369–371. Ramos,A. [2004], Poisson Structures for Reduced Non-Holonomic Systems, J. Phys.A Math. Gen., 37 (2004), 4821–4842. Salamon, S. [1989], Riemannian Geometry and Holonomy Groups, Pitman Research Notes in Mathematics 201, Longman Scientific and Technical, Essex, UK. Schneider, D., Nonholonomic Euler-Poincare equations and stability in Chaplygin’s sphere, Dynam. Systems Intern. J., 17:2, 87–130. Sharpe, R. W. [1997], Differential Geometry: Cartan’s Generalization of Klein’s Erlangen Program, Graduate Texts in Mathematics, Vol. 166, Springer-Verlag, New York, 1997. ´ Sniatycli, J. [1998], Nonholonomic Noether theorem and reduction of symmetries, Rep. Math. Phys., 42:1–2, 5–23.

120


Sn´ iatycki, J. [2001], Almost Poisson spaces and nonholonomic singular reduction, Rep. Math. Phys., 48:1–2, 235–248. ´ Sniatycki, J. [2002], The momentum equation and the second order differential condition, Rep. Math. Phys., 213, 371–394. Sommerfeld, A. [1952], Lectures on Theoretical Physics: Mechanics, Academic Press, New York. Stanchenko, S. V. [1985], Non-holonomic Chaplygin systems, P. M. M. USSR, 53:1, 11–17. Tavares, J. N. [2002], About Cartan Geometrization of Non-Holonomic Mechanics, preprint, Centro de Matemática, Universidade do Porto, Porto, Portugal; available at www.fc.up.pt/cmup. van der Schaft, A., Mashke, B. M. [1994], On the hamiltonian formulation of nonholonomic mechanical systems, Rep. Math. Phys., 34, 225–233. Vaisman, I., Locally conformal symplectic manifolds, Internat. J. Math. Math. Sci., 8:3, 521–536. Vershik, A. M., Gerhskovich, V. [1994], Nonholonomic dynamical systems, geometry of distributions and variational problems, in Arnol’d, V. I., and Novikov, S. P., eds., Dynamical Systems VII, Encyclopedia of Mathematical Sciences, Vol. 16, Springer-Verlag, New York. Vershik, A. M., Fadeev, L. D. [1981], Lagrangian mechanics in invariant form, Selecta Math. Sov., 1:4, 339–350. Veselov, A. P., Veselova, L. E. [1986], Flows on Lie groups with a nonholonomic constraint and integrable non-Hamiltonian systems, Funkt. Anal. Prilozhen., 20:4, 65–66 (in Russian); Functional Anal. Appl., 20:4, 308–309 (in English). Veselov, A. P., Veselova, L. E. [1988], Integrable nonholonomic systems on Lie groups, Mat. Z., 44:5, 604–619, 701 (in Russian); Math. Notes, 44:5–6 (1989), 810–819 (in English). Wade, A. [2000], Conformal Dirac structures, Lett. Math. Phys., 53, 331–348. Warner, F. [1971], Foundations of Differentiable Manifolds and Lie Groups, Scott Foresman, Glenview, IL. Weber, R. W. [1986], Hamiltonian systems with constraints and their meaning in mechanics, Arch. Rational Mech. Anal., 91, 309–335. Whittaker, E. T. [1988], A Treatise on the Analytical Dynamics of Particles and Rigid Bodies, with an Introduction to the Problem of Three Bodies, reprint of the 1937 ed., Cambridge University Press, Cambridge, UK. Zenkov, D. V. [1995], The geometry of the Routh problem, J. Nonlinear Sci., 5:6, 503–519. Zenkov, D. V., Bloch, A. M. [2000], Dynamics of the n-dimensional Suslov problem, J. Geom. Phys., 34:2, 121–136. Zenkov, D. V., Bloch, A. M. [2003], Invariant measures of nonholonomic flows with internal degrees of freedom, Nonlinearity, 16, 1793–1807.

Thompson’s conjecture for real semisimple Lie groups∗ Sam Evens1 and Jiang-Hua Lu2 1 Department of Mathematics

The University of Notre Dame Notre Dame, IN 46556 USA [email protected] 2 Department of Mathematics The University of Hong Kong Pokfulam Road Hong Kong [email protected] Dedicated to Professor Alan Weinstein for his 60th birthday. Abstract. A proof of Thompson’s conjecture for real semisimple Lie groups has been given by Kapovich, Millson, and Leeb. In this paper, we give another proof of the conjecture by using a theorem of Alekseev, Meinrenken, and Woodward from symplectic geometry.

1 Introduction Thompson’s conjecture [T] for the group GL(n, C), which relates eigenvalues of matrix sums and singular values of matrix products, was first proved by Klyachko in [Kl]. In [Al-Me-W], by applying a Moser argument to certain symplectic structures, Alekseev, Meinrenken, and Woodward gave a proof of Thompson’s conjecture for all quasisplit real semisimple Lie groups. In [Ka-Le-M1], Kapovich, Millson, and Leeb have, among other things, proved Thompson’s conjecture for an arbitrary semisimple Lie group G0 . A direct geometric argument can also be found in [Ka-Le-M3, Section 4.2.4]. In this note, we give a different proof of Thompson’s conjecture for arbitrary semisimple real groups by extending the proof of Alekseev, Meinrenken, and Woodward for quasisplit groups. In fact, we prove a stronger result, Theorem 2.2, which implies Thompson’s conjecture. Let G0 = K0 A0 N0 be an Iwasawa decomposition of G0 and let g0 = k0 + p0 be a compatible Cartan decomposition of the Lie algebra of g0 . Theorem 2.2 asserts that for each l ≥ 1, there is a diffeomorphism ∗ The research of the first author was partially supported by NSF grant DMS-9970102. The

research of the second author was partially supported by NSF grant DMS-0105195, by HHY Physical Sciences Fund, and by the New Staff Seeding Fund at HKU.

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S. Evens and J.-H. Lu

L : (A0 N0 )l → (p0 )l which relates the addition on p0 with the multiplication on A0 N0 and intertwines naturally defined K0 -actions. When G0 is quasisplit, Theorem 2.2 follows from results in [Al-Me-W]. The key step in our proof of Theorem 2.2 for an arbitrary G0 is to relate an arbitrary real semisimple Lie algebra g0 to a quasisplit real form in its complexification. In Section 2, we state Theorem 2.2 and show that it implies Thompson’s conjecture. Inner classes of real forms and quasisplit real forms are reviewed in Section 3. The proof of Theorem 2.2 is given in Section 4. Since the version of the Alekseev– Meinrenken–Woodward theorem we present in this paper is not explicitly stated in [Al-Me-W], we give an outline of its proof in Section 5, the appendix.

2 Thompson’s conjecture Let G be a complex connected reductive algebraic group with an antiholomorphic involution τ . Let G0 be a subgroup of the fixed point set Gτ of τ containing the identity connected component. Then G0 is a real reductive Lie group in the sense of [Wa, pp. 42–45], which implies that G0 has Cartan and Iwasawa decompositions. Let g0 be the Lie algebra of G0 . Fix a Cartan decomposition g0 = k0 + p0 of g0 , and let G0 = P0 K0 be the corresponding Cartan decomposition of G0 . Let a0 ⊂ p0 be a maximal abelian subspace of p0 . Fix a choice + res of positive roots in the restricted root system res for (g0 , a0 ), and let n0 be the subspace of g0 spanned by the root vectors for roots in + res . Then g0 = k0 + a0 + n0 is an Iwasawa decomposition for g0 . Let A0 = exp(a0 ) and N0 = exp(n0 ). Then we have the Iwasawa decomposition G0 = K0 A0 N0 for G0 . Consider now the space X0 := G0 /K0 with the left G0 -action given by G0 × (G0 /K0 ) −→ G0 /K0 : (g1 , gK0 ) −→ g1 gK0 ,

g1 , g ∈ G0 .

(2.1)

Thompson’s conjecture is concerned with K0 -orbits in X0 . Identify exp

p0 ∼ = P0 ∼ = G0 /K0 = X0 via the Cartan decomposition G0 = P0 K0 . The K0 -action on X0 in (2.1) becomes the adjoint action of K0 on p0 . Orbits of K0 in p0 are called (real) flag manifolds. Let + a+ 0 ⊂ a0 be the closed Weyl chamber determined by res . It is well known that every + K0 -orbit in p0 goes through a unique element λ ∈ a0 . On the other hand, we can also identify A0 N0 ∼ = G0 /K0 = X0 via the Iwasawa decomposition G0 = A0 N0 K0 . Then the K0 -action on X0 becomes the following action of K0 on A0 N0 : k · b := p(kb) = p(kbk −1 )

for k ∈ K0 , b ∈ A0 N0 ,

(2.2)

Thompson’s conjecture for real semisimple Lie groups

123

where p : G0 → A0 N0 is the projection b1 k1 → b1 for k1 ∈ K0 and b1 ∈ A0 N0 . Let E0 : p0 → A0 N0 be the composition of the identifications: exp

E0 : p0 ∼ = P0 ∼ = G0 /K0 ∼ = A0 N0 .

(2.3)

Then E0 is K0 -equivariant, and E0 (a0 ) = A0 . Thus every K0 -orbit in A0 N0 goes + through a unique point a = exp λ ∈ A+ 0 := exp a0 . Thompson’s conjecture for G0 is concerned with the sum of K0 -orbits in p0 and the product of K0 -orbits in A0 N0 . To further prepare for the statement of the conjecture, let l ≥ 1 be an integer, and consider the two maps a : p0 × p0 × · · · × p0 −→ p0 : (ξ1 , ξ2 , . . . , ξl ) −→ ξ1 + ξ2 + · · · + ξl , m : A0 N0 × A0 N0 × · · · × A0 N0 −→ A0 N0 : (b1 , b2 , . . . , bl ) −→ b1 b2 · · · bl . Clearly, a is K0 -equivariant for the diagonal action of K0 on (p0 )l . On the other hand, define the twisted diagonal action T of K0 on (A0 N0 )l by k −→ Tk := ν −1 ◦ δk ◦ ν : (A0 N0 )l −→ (A0 N0 )l ,

(2.4)

where δk is the diagonal action of k ∈ K0 on (A0 N0 )l , and ν : (A0 N0 )l −→ (A0 N0 )l is the diffeomorphism given by ν(b1 , b2 , . . . , bl ) −→ (b1 , b1 b2 , . . . , b1 b2 · · · bl ).

(2.5)

Them m is K0 -equivariant. See Remark 2.4 for motivation of the twisted diagonal action. Let e be the identity element of A0 N0 and identify Te (A0 N0 ) ∼ = = a0 + n0 ∼ g0 /k0 ∼ . We will regard the map a, respectively, the diagonal K -action on (p0 )l , p = 0 0 as the linearization of the map m, respectively, the twisted diagonal K0 -action on (A0 N0 )l , at the point (e, e, . . . , e). Notation 2.1. For λ ∈ a0 , we will use Oλ to denote the K0 -orbit in p0 through λ. For a ∈ A0 , we will use Da to denote the K0 -orbit in A0 N0 through the point a. If = (λ1 , λ2 , . . . , λl ) ∈ (a0 )l , we set aj = exp(λj ) for 1 ≤ j ≤ l and O = Oλ1 × Oλ2 × · · · × Oλl

and

D = Da1 × Da2 × · · · × Dal .

In this paper, we will prove the following theorem. Theorem 2.2. For every integer l ≥ 1, there is a K0 -equivariant diffeomorphism L : (A0 N0 )l → (p0 )l such that m = E0 ◦ a ◦ L and L(D ) = O for every ∈ (a0 )l . Theorem 2.2 now readily implies the following Thompson’s conjecture for G0 . Corollary 2.3 (Thompson’s conjecture). For each = (λ1 , λ2 , . . . , λl ) ∈ (a0 )l , the two spaces (m−1 (e) ∩ D )/K0 = {(b1 , b2 , . . . , bl ) ∈ D : b1 b2 · · · bl = e}/K0

124


and (a−1 (0) ∩ O )/K0 = {(ξ1 , ξ2 , . . . , ξl ) ∈ O : ξ1 + ξ2 + · · · + ξl = 0}/K0 are homeomorphic. In particular, one is nonempty if and only if the other is. Proof. Let L : (A0 N0 )l → (p0 )l be the diffeomorphism in Theorem 2.2. Then L induces a homeomorphism L : m−1 (e) → a−1 (0). Since L(D ) = O and L is K0 -equivariant, it induces a homeomorphism from (m−1 (e) ∩ D )/K0 to (a−1 (0) ∩ O )/K0 .

Remark 2.4. Equip X0 = G0 /K0 with the G0 -invariant Riemannian structure defined by the restriction of the Killing form of g0 on p0 . For x1 , x2 ∈ X0 , let x1 x2 be the unique geodesic in X0 connecting x1 and x2 . Then there is a unique λ ∈ a+ 0 such that g · x1 = ∗ and g · x2 = (exp λ) · ∗ for some g ∈ G0 , where ∗ = eK0 ∈ X0 is the base + point. The element λ ∈ a+ 0 is called [Ku-Le-M] the a0 -length of x1 x2 . Representing the vertices of an ∗-based l-gon in X0 by (∗, b1 · ∗, b1 b2 · ∗, . . . , b1 b2 · · · bl · ∗) for some b1 , b2 , . . . , bl ∈ A0 N0 , we can regard (b1 , b2 , . . . , bl ) as the set of edges of l the l-gon. Then for ∈ (a+ 0 ) , the space {(b1 , b2 , . . . , bl ) ∈ D : b1 b2 · · · bl = e}/K0 can be identified with the space of G0 -equivalence classes of closed l-gons in X0 with fixed “side length’’ . Similarly, the space {(ξ1 , ξ2 , . . . , ξl ) ∈ O : ξ1 + ξ2 + · · · + ξl = 0}/K0 can be identified with the space of equivalent l-gons with fixed side length in the “infinitesimal symmetric space’’ p0 . Using the right A0 N0 -action on K0 given by k b := q(kb),

b ∈ A0 N0 ,

k ∈ K0 ,

(2.6)

where q : G0 → K0 is the projection q(b1 k1 ) = k1 for b1 ∈ A0 N0 and k1 ∈ K0 , it is easy to see that Tk as defined in 2.4 is also given by Tk (b1 , b2 , . . . , bl ) := (k1 · b1 , k2 · b2 , . . . , kl · bl ),

(2.7)

k b1 b2 ···bj −1

where k1 = k, kj = for 2 ≤ j ≤ l. In the appendix (Section 5), we will see that this formula naturally arises in the context of Poisson Lie group actions. Remark 2.5. When G0 = GL(n,& R), recall that the singular values of g ∈ G0 are by definition the eigenvalues of gg t . Thompson’s conjecture for GL(n, R) says that, for any collection (λ1 , λ2 , . . . , λl ) of real diagonal matrices, the following two statements are equivalent (see [Al-Me-W, Section 4.2]): 1. there exist matrices gj ∈ GL(n, R) whose singular values are entries of aj = exp(λj ) and g1 g2 · · · gl = e; 2. there exist symmetric matrices ξj whose eigenvalues are entries of λj and such that ξ1 + ξ2 + · · · + ξl = 0.


125

Remark 2.6. By a theorem of O’Shea and Sjamaar [O-S], the set a−1 (0) ∩ O is nonempty if and only if = (λ1 , λ2 , . . . , λl ) lies in a certain polyhedral cone P in + l + (a+ 0 ) . For G0 = SL(2, R), we have a0 = R = {λ ∈ R : λ ≥ 0}. In this case 2 p0 may be identified with R and the K0 -action may be identified with rotation. We know from classical triangle inequalities that P for l = 3 is given by the inequalities |λ1 − λ2 | ≤ λ3 ≤ λ1 + λ2 .

(2.8)

The fact that these triangle inequalities are also the necessary and sufficient conditions for λ1 , λ2 and λ3 to be the sides of a geodesic triangle in the hyperbolic 2-space SL(2, R)/SO(2) follows from the law of cosines in this space, which says that cos θ =

cosh λ1 cosh λ2 − cosh λ3 , sinh λ1 sinh λ2

where θ is the angle between the two sides with lengths λ1 and λ2 . For any arbitrary real semisimple Lie group G0 , there have been intensive research activities on the inequalities that describe the polyhedral cone P. We refer to [Ku-Le-M] for explicit examples of these polyhedral cones when X0 has rank 3 and to [Fu, Ka-Le-M1, Ka-Le-M2, Ka-Le-M3] for an account of the history and connections between this problem and others fields such as Schubert calculus, representation theory, symmetric spaces, geometric invariant theory, and integrable systems. See also Remark 4.9. Remark 2.7. Finally, we remark that it is enough to prove Theorem 2.2 for G with trivial center. Indeed, let Z be the center of G, let Z0 = G0 ∩ Z, and let G 0 = G0 /Z0 with Lie algebra g 0 = g0 /z0 , where the Lie algebra z0 of Z0 is the center of g0 . Let j : G0 → G 0 and g0 → g 0 be the natural projections. Let k 0 = j (k0 ) and p 0 = j (p0 ), and let K0 = j (K0 ), A 0 = j (A0 ), and N0 = j (N0 ). By [Kn1, Corollary 1.3], Z0 = (K0 ∩ Z0 )(A0 ∩ Z0 ), and exp : z0 ∩ a0 → Z0 ∩ A0 is an isomorphism. Thus G 0 = K0 A 0 N0 is an Iwasawa decomposition for G 0 , and g 0 = k 0 + p 0 is a Cartan decomposition for g 0 . Moreover, p0 ∼ = p 0 ⊕ (a0 ∩ z0 ) and A0 ∼ = A 0 × (A0 ∩ Z0 ) and ∼ N0 = N0 . Let a : (p 0 )l −→ p 0 ,

m : (A 0 N0 )l −→ A0 N0 ,

a : (a0 ∩ z0 )l −→ a0 ∩ z0 ,

m : (A0 ∩ Z0 )l −→ A0 ∩ Z0

be, respectively, the addition and multiplication maps. If L : (A 0 N0 )l → (p 0 )l is a diffeomorphism satisfying the requirements in Theorem 2.2 for the group G 0 , then L = (L , (log)l ) will be a diffeomorphism from (A0 N0 )l to (p0 )l satisfying the requirements in Theorem 2.2 for the group G0 , where we use the obvious identifications between (A0 N0 )l ∼ = (A 0 N0 )l × (A0 ∩ Z0 )l and (p0 )l ∼ = (p 0 )l × (a0 ∩ z0 )l .

3 Inner classes of real forms and quasisplit real forms Let g be a semisimple complex Lie algebra. Recall that real forms of g are in one-toone correspondence with complex conjugate linear involutive automorphisms of g.

126


For such an involution τ , the corresponding real form is the fixed point set gτ of τ . We will refer to both gτ and τ as the real form. Throughout this paper, if V is a set and σ in an involution on V , we will use V σ to denote the set of σ -fixed points in V . Let G be the adjoint group of g. Definition 3.1 ([A-B-V, Definitions 2.4 and 2.6]). Two real forms τ1 and τ2 of g are said to be inner to each other if there exists g ∈ G such that τ1 = Ad g τ2 . A real form τ of g is said to be quasisplit if there exists a Borel subalgebra b of g such that τ (b) = b. Inner classes of real forms are classified by involutive automorphisms of the Dynkin diagram D(g) of g. Indeed, let Aut g be the group of complex linear automorphisms of g. Its identity component is the adjoint group G. Let Aut D(g) be the automorphism group of the Dynkin diagram D(g) of g. There is a split short exact sequence [A-B-V, Proposition 2.11], !

1 −→ G −→ Aut g −→ Aut D(g) −→ 1.

(3.1)

Denote by R the set of all real forms of g. Let θ be any compact real form of g. Define " : R −→ Aut D(g) : " (τ ) = !(τ θ).

(3.2)

Then " (τ )2 = 1 for each τ , and τ1 and τ2 are inner to each other if and only if " (τ1 ) = " (τ2 ). Conversely, for every involutive d ∈ Aut D(g) , we can construct γd ∈ Aut g such that τ := γd θ is a real form with " (τ ) = d (see (3.4) below). Thus the map " gives a bijection between inner classes of real forms of g and involutive elements in Aut D(g) [A-B-V, Proposition 2.12]). Definition 3.2. Let d be an involutive automorphism of the Dynkin diagram D(g) of g. We say that a real form τ of g is of inner class d or in the d-inner class if " (τ ) = d. By [A-B-V, Proposition 2.7], every inner class of real forms of g contains a quasisplit real form that is unique up to G-conjugacy. In the following, for each involutive d ∈ Aut D(g) , we will construct an explicit quasisplit real form τd in the d-inner class. We will then show that, up to G-conjugacy, every real form in the d-inner class is of the form τ = Ad w˙ 0 τd , where w0 is a certain Weyl group element and w˙ 0 a representative of w0 in G. We first fix once and for all the following data for g: Let h be a Cartan subalgebra of g, and let be the corresponding root system. Fix a choice of positive roots + in , and let be the basis of simple roots. Let ·, · be the Killing form on g. For each α ∈ , let E±α be root vectors such that [Eα , E−α ] = Hα for all α ∈ + , where Hα is the unique element of h defined by H, Hα = α(H ) for all H ∈ h, and the numbers mα,β for α, β ∈ defined for α = −β by [Eα , Eβ ] = mα,β Eα+β =0

if α + β ∈ otherwise


127

satisfy m−α,−β = −mα,β . We will refer to the set {Eα , E−α : α ∈ + } as (part of) a Weyl basis. Using a Weyl basis {Eα , E−α : α ∈ + }, we can define a compact real form k of g as √ √ k = spanR { −1Hα , Xα := Eα − E−α , Yα := −1(Eα + E−α ) : α ∈ + }. (3.3) Let θ be the complex conjugation of g defining k. We also define a split real form η0 of g by setting η0 |a = id, and η0 (Eα ) = Eα for every α ∈ . Clearly θ η0 = η0 θ. The inner class for η0 is easily seen to be the automorphism of the simple roots given by −w 0 , where w 0 is the longest element in the Weyl group W of (g, h). An explicit splitting of the short exact sequence (3.1) can be constructed using the Weyl basis. Indeed, for any d ∈ Aut D(g) , define γd ∈ Aut g by requiring γd (Hα ) = Hdα

and

γd (Eα ) = Edα

(3.4)

for each simple root α. Then d → γd is a group homomorphism from Aut D(g) to Aut g and is a section of ! in (3.1). Moreover, every γd commutes with both θ and η0 because they commute on a set of generators of g. Lemma 3.3. For an involutive element d ∈ Aut D(g) , let γ−w0 d ∈ Aut g be the lifting of −w0 d ∈ Aut D(g) as defined in (3.4). Define τd = η0 γ−w0 d .

(3.5)

Then τd is a quasisplit real form of g in the d-inner class. Proof. We know that (τd )2 = 1 because −w0 ∈ Aut D(g) is in the center. Since τd maps every positive root vector to another positive root vector, it is a quasisplit real form. Finally, since " (τd ) = !((γ−w0 )(γ−w0 d )) = d, we see that τd is in the d-inner class.

To relate an arbitrary real form in the d-inner class with the quasisplit real form = k + a + n is an Iwasawa τd , we recall some definitions from [Ar]. Note first that g decomposition, where a = spanR {Hα : α ∈ } and n = α∈ + gα . Definition 3.4. A real form τ of g is said to be normally related to (k, a) and compatible with + if 1. τ θ = θ√ τ , and τ (h) = h; √ 2. aτ ⊂ ( −1k)τ is maximal abelian in ( −1k)τ ; 3. if α ∈ + is such that α|aτ = 0, then τ (α) ∈ + , where τ (α) ∈ a∗ is defined by τ (α)(λ) = α(τ (λ)) for λ ∈ a. We will call a real form with properties 1–3 an Iwasawa real form relative to (k, a, n). Remark 3.5. Once properties 1 and 2 in Definition 3.4 are satisfied, property 3 is equivalent to the set r( + )\{0} ⊂ res being a choice of positive roots for the restricted root system res of (gτ , aτ ), where r is the map dual to the inclusion aτ → a. If τ is an Iwasawa real form relative to (k, a, n), then so is Ad t τ Ad −1 t for any t ∈ exp(ia).

128


Proposition 3.6. 1. Every real form of g is conjugate by an element in G to a real form that is Iwasawa relative to (k, a, n). 2. Suppose that τ is an Iwasawa real form relative to (k, a, n) and suppose that τ is in the d-inner class. Let w0 be the longest element of the subgroup of W generated by the reflections corresponding to roots in the set 0

= {α ∈

: α|aτ = 0} = {α ∈

: τ (α) = −α}.

Then there is a representative w˙ 0 of w0 in G such that τ = Ad w˙ 0 τd .

(3.6)

Proof. Statement 1 follows from [Ar, Proposition 1.2, Section 2.8, and Corollary 2.5]. Statement 2: Assume now that τ is an Iwasawa real form relative to (k, a, n) and that τ is in the d-inner class. Consider τd τ . Since both τ and τd are in the d-inner class, τd τ = Ad g for some g ∈ G. Since both τ and τd leave h invariant, the element g represents an element in the Weyl group W . Let 0 = ∩ 0 . By [Ar, Section 2.8], α ∈ 0 if and only if α is in the linear span of 0 . For every α ∈ 0 , we have τd τ (α) = −τd (α) ∈ − + , and for every α ∈ + − 0 , since τ (α) ∈ + , we have

(τd τ )(α) ∈ + . Thus g represents the element w0 = (w0 )−1 . Remark 3.7. Recall from [Ar] that the Satake diagram of τ is the Dynkin diagram of g with simple roots in 0 painted black, simple roots in − 0 painted white, and a two-sided arrow drawn between two white simple roots α and α if τ (α) = α + β for some β ∈ 0 . From (3.6) we see that α = −w0 d(α) if α is a white simple root. Conversely, given a Satake diagram for a real form of g, let c ∈ Aut D(g) be defined by + −w0 α if α is black, (3.7) c(α) = if α is white, α where w0 is the longest element in the subgroup of the Weyl group of (g, h) generated by the black dots in the Satake diagram, and α → α is the order-2 involution on the set of white dots in the diagram. Then c is involutive, and the inner class of the real form is d = −w0 c. We now return to the real form τ in Proposition 3.6. Set + 1

= {α ∈

Then τ (

+ 1)

⊂

+

: α|aτ = 0},

+ 1.

(

+ 1)

=

+

∩

0

= {α ∈

+

: α|aτ = 0}.

Set n1 =

α∈

+ 1

gα ,

n 1 =

α∈(

gα .

(3.8)

+ 1)

Then n1 is τ -invariant, and, since there are no noncompact imaginary roots for the Cartan subalgebra hτ of gτ , we have τ |n 1 = θ|n 1 [Ar, Proposition 1.1]. Since the


restriction of know that

+

129

to aτ gives a choice of positive restricted roots for (gτ , aτ ), we gτ = kτ + aτ + (n1 )τ

is an Iwasawa decomposition of

(3.9)

gτ .

4 Proof of Theorem 2.2 By Remark 2.7, it is enough to prove Theorem 2.2 when G of adjoint type. Let g0 be a real form of g, the Lie algebra of G. Then by Proposition 3.6, we can assume that g0 = gτ , where τ is the involution on g given by (3.6), and d is the inner class of g0 . The lifting of τ to G will also be denoted by τ . Let G0 contain the connected component of the identity of the subgroup Gτ . In this section, we will prove Theorem 2.2 for G0 . The first step in our proof of Theorem 2.2 for G0 is to realize the various objects associated to G0 as fixed point sets of involutions on the corresponding objects related to G. We will then apply a theorem of Alekseev–Meinrenken–Woodward, stated as Theorem 4.7 below, whose proof using Poisson geometry will be outlined in Section 5, the appendix. We will keep all the notation from Section 3. In particular, set √ k0 = kτ , p0 = ( −1k)τ , a0 = aτ , and n0 = (n1 )τ . Then g0 = k0 +p0 is a Cartan decomposition of g0 , and g0 = k0 +a0 +n0 an Iwasawa decomposition of g0 . Let K be the connected subgroup of G with Lie algebra k. Let K0 = K ∩ G0 , K τ = K ∩ Gτ , and let N1 = exp(n1 ),

A0 = exp(a0 ),

and

N0 = N1 ∩ Gτ = exp(n0 ).

Lemma 4.1. G0 = K0 A0 N0 is an Iwasawa decomposition of G0 , and Gτ = K τ A0 N0 is an Iwasawa decomposition of Gτ . Proof. The statements follow from [Wa, Lemma 2.1.7] and the facts that K0 and K τ are maximally compact subgroups of G0 and of Gτ, respectively.

Let A = exp a and N = exp n so that G = KAN is an Iwasawa decomposition of G. We will now identify A0 N0 with the fixed point set of an involution on AN, although we note that the involution τ does not leave AN invariant unless τ = τd . Define σ : AN −→ AN : σ (b) = p(τ (b)), (4.1) where p : G = KAN → AN is the projection b1 k1 → b1 for k1 ∈ K and b1 ∈ AN. Recall from (3.6) that τ = Ad w˙ 0 τd on g. Since both τ and τd commute with θ, the element w˙ 0 is in K. As for the case of G0 , we can use the Iwasawa decomposition G = KAN to define a left action of K on AN ∼ = G/K by k · b := p(kb),

k ∈ K,

b ∈ AN.

(4.2)

130


Then σ : AN → AN is also given by σ (b) = w˙ 0 · τd (b)

for b ∈ AN .

(4.3)

Lemma 4.2. σ : AN → AN is an involution, and A0 N0 = (AN )σ , the fixed point set of σ in AN. Proof. The fact that σ 2 = 1 follows from the fact that w˙ 0 τd (w˙ 0 ) = 1. Recall that A0 N0 is the fixed point set of τ in AN1 , where N1 = exp(n1 ) and n1 ⊂ n is given in (3.8). Since σ coincides with τ on AN1 , we have A0 N0 ⊂ (AN )σ . Suppose now that b ∈ AN is such that σ (b) = b. Then there exists k ∈ K such that τ (b) = bk. By [Sl, Proposition 7.1.3], we can decompose b as b = gak1 for some k1 ∈ K, a ∈ A and g ∈ Gτ . Then τ (b) = gτ (a)τ (k1 ), and thus gτ (a)τ (k1 ) = gak1 k, from which it follows that τ (a) = a and τ (k1 ) = k1 k. Thus k = k1−1 τ (k1 ), and hence τ (bk1−1 ) = bk1−1 . Write bk1−1 = b2 k2 with k2 ∈ K τ and b2 ∈ A0 N0 using the Iwasawa decomposition of Gτ . It follows then that k2 = k1−1 and b2 = b, so b ∈ A0 N0 .

Now let l ≥ 1 be an integer. As in Section 2, we have the twisted diagonal action k → Tk of K on (AN )l given by Tk = ν −1 ◦ δk ◦ ν : (AN )l −→ (AN )l ,

(4.4)

where ν : (AN )l → (AN )l is as in (2.5) with A0 N0 replaced by AN, and δk denotes the diagonal action of k ∈ K on AN. Set (τd )l = (τd , τd , . . . , τd ) : (AN )l → (AN )l . Lemma 4.3. For an integer l ≥ 1, define σ (l) = Tw˙ 0 ◦ (τd )l : (AN )l −→ (AN )l . Then σ (l) is an involution, and the fixed point set of σ (l) is (A0 N0 )l . Proof. Let σ l = (σ, σ, . . . , σ ) : (AN )l → (AN )l , where σ : AN → AN is as in Lemma 4.2. Since τd is a group automorphism of AN, we have σ (l) = ν −1 ◦ δw˙ 0 ◦ ν ◦ (τd )l = ν −1 ◦ (δw˙ 0 ◦ (τd )l ) ◦ ν = ν −1 ◦ σ l ◦ ν. Thus (σ (l) )2 = 1. Moreover, let b = (b1 , b2 , . . . , bl ) ∈ (AN )l , and let b = ν(b). Then σ (l) (b) = b if and only if σ l (b ) = b , which in turn is equivalent to bj ∈ A0 N0 for each 1 ≤ j ≤ l because of Lemma 4.2 and because of the fact that A0 N0 is a subgroup of AN.

√ Let p = −1k, so g = k + p is a Cartan decomposition of g. Let E : p → AN be the composition of the identifications exp

E:p ∼ = exp(p) ∼ = G/K ∼ = AN.

(4.5)

Then E is K-equivariant with respect to the action of K on p by conjugation and the action of K on AN given in (4.2).


131

Lemma 4.4. E ◦ (τ |p ) = σ ◦ E, and E0 = E|p0 : p0 → A0 N0 . Proof. Consider E −1 : AN → p. For g ∈ G, define g ∗ = θ (g −1 ). Then for every b ∈ AN, E −1 (b) = 12 log(bb∗ ) for all b ∈ AN, and thus 1 log(w˙ 0 τd (b)τd (b)∗ w˙ 0−1 ) 2 1 log(τd (b)τd (b)∗ ) = Ad w˙ 0 τd (E −1 (b)) = τ (E −1 (b)). = Ad w˙ 0 2

E −1 (σ (b)) =

Thus E ◦ (τ |p ) = σ ◦ E, and E(p0 ) = A0 N0 by Lemma 4.2. It also follows that E|p0 = E0 .

Notation 4.5. For λ ∈ a ⊂ p, let Oλ be the K-orbit in p through λ, and let Da be the K-orbit in AN through a = exp λ ∈ A. For = (λ1 , λ2 , . . . , λl ) ∈ (a)l , set O = Oλ1 × Oλ2 × · · · × Oλl

and

D = Da1 × Da2 × · · · × Dal .

(4.6)

Recall from Section 2 that, for λ ∈ a0 , Oλ denotes the K0 -orbit in p0 through λ, and Da denotes the K0 -orbit in A0 N0 through a = exp λ ∈ A0 . Lemma 4.6. Let λ ∈ a0 and a = exp λ ∈ A0 . Then 1. τd (λ) = λ, so both Oλ ⊂ p and Da ⊂ AN are τd -invariant; 2. Oλ is τ -invariant, and (Oλ )τ = Oλ ; 3. Da is σ -invariant and (Da )σ = Da . Proof. 1. Let α be a simple root such that τ (α) = −α. Then for any λ ∈ a0 , α(λ) = α(τ (λ)) = (τ (α))(λ) = −α(λ) = 0. Thus rα (λ) = λ, where rα is the reflection in a defined by α. Since w0 is a product of such reflections (see Proposition 3.6), we see that w0 acts trivially on a0 . Thus every λ ∈ a0 is also fixed by τd . 2. This is a standard fact. See, for example, [O-S, Example 2.9]. We remark that the key point is to show that (Oλ )τ is connected. 3. Statement 3 follows from statement 2 and Lemma 4.4.

We can now state the Alekseev–Meinrenken–Woodward theorem. Set a : p × p × · · · × p −→ p : (x1 , x2 , . . . , xl ) −→ x1 + · · · + xl , m : AN × AN × · · · × AN −→ AN : (b1 , b2 , . . . , bl ) −→ b1 b2 · · · bl . As for the case of G0 , we will equip pl with the diagonal K-action by conjugation, and we will equip (AN )l with the twisted diagonal action T given by (4.4).

132


Theorem 4.7 (Alekseev–Meinrenken–Woodward [Al-Me-W]). For every quasisplit real form τd given in (3.5) and for every integer l ≥ 1, there is a K-equivariant diffeomorphism L : (AN )l → pl such that m = E ◦ a ◦ L,

and (τd )l ◦ L = L ◦ (τd )l .

Moreover, L(D ) = O for every ∈

(4.7)

al .

Remark 4.8. Theorem 4.7, whose proof will be outlined in the appendix (Section 5), is a consequence of the Moser isotopy lemma for Hamiltonian K-actions on Poisson manifolds, a rigidity theorem for such spaces. More precisely, we will see in the appendix (Section 5) that the map E −1 ◦ m : (AN )l → p is a moment map for the twisted diagonal K-action T on (AN )l with respect to a Poisson structure π1 on (AN)l , and (τd )l is an anti-Poisson involution for π1 . Moreover, the symplectic leaves of π1 are precisely all the orbits O for ∈ al . The quintuple Q1 = ((AN )l , π1 , T , E −1 ◦ m, (τd )l ) will be referred to as a Hamiltonian Poisson K-space with anti-Poisson involution. In fact, Q1 belongs to a smooth family Qs = ((AN )l , πs , Ts , E −1 ◦ ms , (τd )l ) as the case for s = 1, and when s = 0, Ts is the diagonal K-action on (AN )l and E −1 ◦ m0 = a ◦ (E −1 )l . The Moser isotopy lemma, Proposition 5.1 in Section 5, implies that Qs is isomorphic to Q0 by a diffeomorphism ψs of (AN )l for every s ∈ R. The map L in Theorem 4.7 is then taken to be (E −1 )l ◦ ψ1 . We will assume Theorem 4.7 for now and prove Theorem 2.2 for G0 . Proof of Theorem 2.2. Let L : (AN )l → pl be as in Theorem 4.7. Since L is Kequivariant and intertwines (τd )l : (AN )l → (AN )l and (τd )l : pl → pl , it also intertwines σ (l) = Tw˙ 0 ◦ (τd )l : (AN )l −→ (AN )l

and

τ l = δw˙ 0 ◦ (τd )l : pl −→ pl .

Thus by Lemma 4.3, we know that L((A0 N0 )l ) = (p0 )l . Denote L|(A0 N0 )l : (A0 N0 )l → (p0 )l also by L. Then clearly L is K0 -equivariant, and since E0 : p0 → A0 N0 coincides with the restriction of E : p → AN to p0 , we see that m = E0 ◦a ◦L. Finally, let = (λ1 , λ2 , . . . , λl ) ∈ (a0 )l . Then by Lemma 4.6, we see that L(D ) = L(D ∩ (A0 N0 )l ) = O ∩ (p0 )l = O .

+ Remark 4.9. Let a+ = {x ∈ a : α(x) ≥ 0 ∀α ∈ + } so that a+ 0 = a0 ∩ a . By + l Kirwan’s convexity theorem, there exists a polyhedral cone P ⊂ (a ) such that ∈ P if and only if a−1 (0) ∩ O is nonempty. The cone P is explicitly computed l in [B-S]. Set P0 = P ∩ (a0 )l ⊂ (a+ 0 ) . Then by a theorem of O’Shea–Sjamaar [O-S], −1 the set a (0) ∩ O is nonempty if and only if ∈ P0 . If we use Pd ⊂ (aτd )l to denote the polyhedral cone P ∩ (aτd )l for the quasisplit form τd , it follows from a0 ⊂ aτd that P0 = Pd ∩ (a0 )l . (4.8)

A statement related to this fact is given in [Fo].


133

5 Appendix: Alekseev–Meinrenken–Woodward theorem In this appendix, we give an outline of the proof of the Alekseev–Meinrenken– Woodward theorem, stated as Theorem 4.7 in this paper. [Al-Me-W, Theorem 3.5] shows the existence of a diffeomorphism L : D → O satisfying (4.7) for each ∈ al . To show that all the L ’s come from a globally defined L on all of (AN)l , one uses the Moser isotopy lemma for Hamiltonian Poisson Kspaces proved in [Al-Me]. What we present here is a collection of arguments from [Al, Al-Me-W, Ka-M-T, Al-Me]. 5.1 Gauge transformation for Poisson structures Recall that a Poisson structure on a manifold M is a smooth section π of ∧2 T M such that [π, π] = 0, where [ , ] is the Schouten bracket on the space of multi-vector fields on M. For a smooth section π of ∧2 T M, we will use π # to denote the bundle map π # : T ∗ M → T M : π # (α) = π(·, α) for all cotangent vectors α. Similarly, for a 2-form γ on M, we will set γ # : T M → T ∗ M : γ # (v) = γ (·, v) for all tangent vectors v. Suppose now that π is a Poisson structure on M and that γ is a closed 2-form on M. If the bundle map 1 + γ # π # : T ∗ M → T ∗ M is invertible, the section π of ∧2 T M given by (π )# = π # (1 + γ # π # )−1 : T ∗ M −→ T M

(5.1)

is then a Poisson structure on M. The Poisson structure π will be called the gauge transformation of π by the closed 2-from γ , and we write π = Gγ (π ). It is clear from (5.1) that π and π have the same symplectic leaves. If S is a common symplectic leaf, then the symplectic 2-forms ω and ω coming from π and π differ by iS∗ γ , where iS : S → M is the inclusion map. See [Se-W] for more details. 5.2 The Poisson Lie groups (K, sπK ) and (AN, •s , πAN,s ) The group AN carries a distinguished Poisson structure πAN . Indeed, let , be the imaginary part of the Killing form of g and identify k with (a + n)∗ via , . For x ∈ k, denote by x¯ the right-invariant 1-form on AN defined by x. Let xAN be the generator of the action of exp(tx) on AN according to (4.2). Then the unique section πAN of ∧2 T (AN) such that # (x) ¯ = xAN ∀x ∈ k πAN (5.2) is a Poisson bivector field on AN. The Poisson structure πAN makes AN into a Poisson Lie group in the sense that the group multiplication map AN × AN → AN : (b1 , b2 ) → b1 b2 is a Poisson map, where AN × AN is equipped with the product Poisson structure πAN × πAN . We refer to [L-W] and [L] for details on Poisson Lie groups and Poisson Lie group actions and to [L-Ra]) for details on πAN . In particular, the dual Poisson Lie group of (AN, πAN ) is K together with the Poisson structure πK , explicitly given by πK = r0 − l0 , where

134


0 =

1 Xα ∧ Yα ∈ ∧2 k 2 + α∈

with Xα , Yα ∈ k given in (3.3) and r0 and l0 being, respectively, the right- and left-invariant bivector fields on K determined by 0 . It follows from (5.2) that the symplectic leaves of πAN are precisely the orbits of the K-action on AN given in (4.2). Now let d be an involutive automorphism of the Dynkin diagram of g, and let τd be the quasisplit real form of g given in (3.5). Recall that τd leaves AN invariant and defines a group isomorphism on AN. It is easy to check (see also [Al-Me-W, Section 2.3]) that τd : (AN, πAN ) → (AN, πAN ) is anti-Poisson, i.e., τd ∗ πAN = −πAN . Similarly, τd : K → K is anti-Poisson for πK . We will denote the restrictions of τd to K and to AN both by τd , and we will refer to (K, πK , τd ) and (AN, πAN , τd ) as a dual pair of Poisson Lie groups with anti-Poisson involutions. In the context of Poisson Lie groups, the K-action on AN given in (4.2) and the AN-action on K given in (2.6) (with AN replacing A0 N0 and K replacing K0 ) are, respectively, called the dressing actions. As noticed in [Al] and [Ka-M-T], we in fact have a smooth family of Poisson Lie groups (AN, •s , πAN,s ) for s ∈ R. Indeed, for s ∈ R − {0}, let Fs : p → p be the diffeomorphism x → sx, and let Is = E ◦ Fs ◦ E −1 : AN → AN. Let πAN,s be the Poisson bivector field on AN such that (Is )∗ πAN,s = sπAN , or πAN,s (b) = s(Is−1 )∗ (πAN (Is (b))),

b ∈ AN.

(5.3)

Define the group structure •s : AN × AN → AN by b1 •s b2 := Is−1 (Is (b1 )Is (b2 )),

b1 , b2 ∈ AN.

Then since s = 0, the map (AN ×AN, πAN,s ×πAN,s ) → (AN, πAN,s ) : (b1 , b2 ) → b1 b2 is a Poisson map, so (AN, •s , πAN,s ) is a Poisson Lie group for each s ∈ R, s = 0. On the other hand, p ∼ = k∗ has the linear Poisson structure πp,0 defined by the Lie algebra k. Let •0 and let πAN,0 be the pullbacks to AN by E −1 : AN → p of the abelian group structure on p and the Poisson structure πp,0 on p. Then we get a smooth family of Poisson Lie group structures (•s , πAN,s ) on AN for every s ∈ R (see [Al] and [Ka-M-T]). The dual Poisson Lie group of (AN, •s , πAN,s ) is again the Lie group K (with group structure independent on s) but with the Poisson structure sπK , if we identify again k ∼ = (a + n)∗ via the imaginary part of the Killing form of g. It is also clear that τd is a group isomorphism for •s and is anti-Poisson for πAN,s . Thus we get a dual pair of Poisson Lie groups (K, sπK , τd ) and (AN, •s , πAN,s , τd ) with anti-Poisson involutions for each s ∈ R. 5.3 The Poisson structure πs on (AN )l As noted in [Al], for each s ∈ R, the Poisson structure πAN,s on AN is related to πAN by a gauge transformation. Recall that for x ∈ k ∼ = (a + n)∗ , x¯ is the right-invariant 1-form on AN defined by x. Let lx be the differential of the linear function ξ → x, ξ


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on p, and let xp be the vector field on p generating the adjoint action of exp(tx) ∈ K on p. By [Al-Me-W, Proposition 3.1], there is a 1-form β on p such that β(0) = 0 and −(dβ)# (xp ) = E ∗ x¯ − lx

∀x ∈ k.

Moreover, (τd )∗ β = −β for every quasisplit real form τd given in (3.5). For s ∈ R − {0}, let βs = 1s (Fs∗ β). Since β(0) = 0, the family βs extends smoothly to β0 = 0. Let 1 α = (E −1 )∗ β and αs = (E −1 )∗ βs = (Is∗ α) s for all s ∈ R. Then it is easy to show that, for every s ∈ R, πAN,s = Gd(α−αs ) (πAN ) = G−dαs (πAN,0 ). Assume now that l ≥ 1 is an integer. For each s ∈ R, set ms : (AN )l −→ AN : (b1 , b2 , . . . , bl ) −→ b1 •s b2 •s · · · •s bl . By generalizing the “linearization" procedure of Hamiltonian symplectic (K, sπK )spaces described in [Al-Me-W] to the case of Poisson manifolds, one can show that πs := Gdms∗ αs (πAN,s × πAN,s × · · · × πAN,s )

(5.4)

is a well-defined Poisson structure on (AN )l for each s ∈ R. Define the twisted diagonal action Ts of K on (AN )l by k −→ Ts,k := νs−1 ◦ δk ◦ νs ,

(5.5)

where, again, δk denotes the diagonal action of k on (AN )l for the action of K on AN given in (4.2), and νs ∈ Diff ((AN )l ) is given by νs (b1 , b2 , . . . , bl ) = (b1 , b1 •s b2 , . . . , b1 •s b2 •s · · · •s bl ). Note that Ts,k is Tk when s = 1 and is δk when s = 0. Then again it follows from [Al-Me-W] that for each s ∈ R, the action Ts of K on (AN )l is Hamiltonian with respect to the Poisson structure πs with the map E −1 ◦ ms : (AN )l → p ∼ = k∗ as a moment map. Moreover, for every quasisplit real form τd defined in (3.5), the Cartesian product (τd )l = τd × τd × · · · × τd is anti-Poisson for πs for every s ∈ R. 5.4 Moser isotopy lemma Let U be a connected Lie group with Lie algebra u. Suppose that σU is an involutive automorphism of U with the corresponding involution on u denoted by σu . Define σu∗ = −(σu )∗ . If (M, πM , ) is a Hamiltonian Poisson U -space, an anti-Poisson involution σM of (M, πM ) is said to be compatible with σU if ◦ σM = σu∗ ◦ . The following Moser isotopy lemma for Hamiltonian Poisson U -spaces with anti-Poisson involutions is proved in [Al-Me]. See [Al-Me-W] for the symplectic case.

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Proposition 5.1. Let U be a connected compact semisimple Lie group with Lie algebra u, and let (M, πs , s ), s ∈ R, be a smooth family of Hamiltonian Poisson U -spaces. Suppose that there exists a smooth family of 1-forms s on M with 0 = 0 such that πs = Gds π0 for every s ∈ R. Assume also that π0 has compact symplectic leaves. Then (M, πs , s ) is isomorphic to (M, π0 , 0 ) for every s ∈ R as Hamiltonian Poisson U -spaces, i.e., there exists ψs ∈ Diff (M) for s ∈ R with ψ0 = id, such that for every s ∈ R, (1) πs = ψs ∗ π0 ; (2) s ◦ ψs = 0 . If σU is an involutive automorphism on U , and if for each s ∈ R, σM,s is an anti∗ ˙ = −˙ s , where Poisson involution for πs compactible with σU and such that σM,s s d ˙s = ds s for s ∈ R, then ψs can be chosen such that ψs ◦ σM,0 = σM,s ◦ ψs for all s ∈ R. 5.5 Proof of Theorem 4.7 Consider the Hamiltonian Poisson K-space (M = (AN )l , πs , s ) with s = E −1 ◦ ms . The action of K on (AN )l induced by (πs , s ) is the twisted diagonal action Ts given in (5.4). From the definition of πs , we know that πs = Gds π0 , where s = ms∗ αs −

l

pj∗ αs

j =1

with pj : (AN )l → AN denoting the projection to the j ’th factor. For every quasisplit real form τd given in (3.5), since τd is a group isomorphism for (AN, •s ), we have τd∗ s = −s , and thus τd∗ ˙s = −˙s for every s ∈ R. Let σM,s = (τd )l and let ψs ∈ Diff ((AN )l ) be as in Proposition 5.1. Then L := (E −1 )l ◦ψ1−1 : (AN )l → (p)l is the diffeomorphism in Theorem 4.7. Indeed, E ◦ a ◦ L = E ◦ a ◦ (E −1 )l ◦ ψ1−1 = E ◦ 0 ◦ ψ1−1 = E ◦ 1 = m, where the second equality follows from the identity a ◦ (E −1 )l = E −1 ◦ m0 , which is a trivial consequence of the fact that m0 is the pullback of addition by the map E.

Acknowledgments Although we do not explicitly use any results from [Fo], our paper is very much inspired by [Fo]. We thank P. Foth for showing us a preliminary version of [Fo] and for helpful discussions. We also thank J. Millson and M. Kapovich for sending us the preprint [Ka-Le-M1] and R. Sjamaar for answering some questions. Thanks also go to the referee for helpful comments.

References [A-B-V]

Adams, J., Barbasch, D., and Vogan, D., The Langlands Classification and Irreducible Characters for Real Reductive Groups, Birkhäuser, Boston, 1992.

Thompson’s conjecture for real semisimple Lie groups [Al] [Al-Me-W]

[Al-Me] [Ar] [B-S] [Fo] [Fu] [Ka-Le-M1] [Ka-Le-M2] [Ka-Le-M3]

[Ka-M-T] [Kl] [Kn1] [Ku-Le-M]

[L-W] [L]

[L-Ra] [O-S] [Sl] [Se-W]

[T] [Wa]

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Alekseev, A., On Poisson actions of compact Lie groups on symplectic manifolds, J. Differential Geom., 45 (1997), 241–256. Alekseev, A., Meinrenken, E., and Woodward, C., Linearization of Poisson actions and singular values of matrix products, Ann. Inst. Fourier Grenoble, 51-6 (2001), 1691–1717. Alekseev, A., and Meinrenken, E., Poisson geometry and the Kashiwara–Vergne conjecture, C. R. Math. Acad. Sci. Paris, 335 (2002), 723–728. Araki, S., On root systems and an infinitesimal classification of irreducible symmetric spaces, J. Math. Osaka City Univ., 13-1 (1962), 1–34. Berenstein, A., and Sjamaar, R., Coadjoint orbits, moment polytopes, and the Hilbert–Mumford criterion, J. Amer. Math. Soc., 13-2 (2000), 433–466. Foth, P., A note on Lagrangian loci of quotients, Canad. Math. Bull., to appear; math.SG/0303322. Fulton, W., Eigenvalues, invariant factors, highest weights, and Schubert calculus, Bull. Amer. Math. Soc. (N.S.), 37-3 (2000), 209–249. Kapovich, M., Leeb, B., and Millson, J., Polygons in symmetric spaces and buildings, preprint, 2002. Kapovich, M., Leeb, B., and Millson, J., The generalized triangle inequalities in symmetric spaces and buildings with applications to algebra, math.RT/0210256. Kapovich, M., Leeb, B., and Millson, J., Convex functions on symmetric spaces and geometric invariant theory for weighted configurations on flag manifolds, math.DG/0311486. Kapovich, M., Millson, J., and Treloar, T., The symplectic geometry of polygons in hyperbolic 3-space, Asian J. Math., 4-1 (2000) (Kodaira’s issue), 123–164. Klyachko, A., Random walks on symmetric spaces and inequalities for matrix spectra, Linear Algebra Appl., 319-1–3 (2000), 37–59. Knapp, A., Representation Theory of Semi-Simple Groups, Princeton University Press, Princeton, NJ, 1986. Kumar, S., Leeb, B., and Millson, J., The generalized triangular inequalities for rank 3 symmetric spaces of non-compact type, in Explorations in Complex and Riemannian Geometry: A Volume Dedicated to Robert Greene, Contemporary Mathematics, Vol. 332, American Mathematical Society, Providence, RI, 2003, 171–195. Lu, J.-H., and Weinstein, A., Poisson Lie groups, dressing transformations, and Bruhat decompositions, J. Differential Geom., 31 (1990), 501–526. Lu, J.-H., Moment mappings and reductions of Poisson Lie groups, in Proc. Seminaire Sud-Rhodanien de Géométrie, Mathematical Sciences Research Institute Publications Series, Springer-Verlag, New York, 1991, 209–226. Lu, J.-H., and Ratiu, T., On the non-linear convexity theorem of Kostant, J. Amer. Math. Soc., 4-2 (1991), 349–361. O’Shea, L., and Sjamaar, R., Moment maps and Riemannian symmetric pairs, Math. Ann., 317-3 (2000), 415–457. Schlichtkrull, H., Hyperfunctions and Harmonic Analysis on Symmetric Spaces, Birkhäuser, Basel, 1984. Severa, P., and Weinstein, A., Poisson geometry with a 3-form background, in Proceedings of the International Workshop on Non-Commutative Geometry and String Theory, Keio University, Tokyo, 2001; also available at math.SG/0107133. Thompson, R., Matrix Spectral Inequalities, John Hopkins University Press, Baltimore, 1988. Wallach, N., Real Reductive Groups I, Academic Press, New York, 1988.

The Weinstein conjecture and theorems of nearby and almost existence∗ Viktor L. Ginzburg Department of Mathematics University of California at Santa Cruz Santa Cruz, CA 95064 USA [email protected] Dedicated to Alan Weinstein on the occasion of his 60th birthday. Abstract. The Weinstein conjecture, as the general existence problem for periodic orbits of Hamiltonian or Reeb flows, has been among the central questions in symplectic topology for over two decades and its investigation has led to understanding some fundamental properties of Hamiltonian flows. In this paper we survey some recently developed and well-known methods of proving various particular cases of this conjecture and the closely related almost existence theorem. We also examine differentiability and continuity properties of the Hofer–Zehnder capacity function and relate these properties to the features of the underlying Hamiltonian dynamics, e.g., to the period growth.

1 Introduction Without exaggeration, one can say that Arnold’s conjecture and the Weinstein conjecture have been the two problems determining the development of symplectic topology over the past twenty years. The Weinstein conjecture [We4], the problem we are interested in here, concerns the existence of closed characteristics on a compact hypersurface of contact type. To be more precise, consider a regular compact contact type level of a Hamiltonian on a symplectic manifold. Then, the Weinstein conjecture as we understand it now asserts that the level must carry at least one periodic orbit of the Hamiltonian flow. This paper is a survey of some recent and well-known results concerning a particular perspective on the Weinstein conjecture, originating from the so-called almost existence theorem. The main focus of this survey is on the action selector and symplectic capacity methods. Arguing along the lines of these methods, we reprove a number ∗ The work is partially supported by the NSF and by the faculty research funds of the University

of California at Santa Cruz.

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of particular cases of the conjecture and also refine the capacity–displacement energy inequality for noncompact convex symplectically aspherical manifolds (see Sections 2.5.2 and 3.3) and analyze in Section 4 the problem of continuity of the Hofer–Zehnder capacity. Some aspects of the conjecture are just touched upon or not considered at all in this survey. Among the latter is, for instance, the Weinstein conjecture for general contact manifolds. The contents of the survey are outlined in more detail at the end of the introduction. The Weinstein conjecture was motivated by numerous results establishing the existence of periodic orbits under various, often rather restrictive, conditions on the level (e.g., convex or bounding a star-shaped domain); see, e.g., [Mo, Ra, We1, We2, We3]. The feature distinguishing the Weinstein conjecture from these results is the requirement that the level have contact type is invariant under symplectomorphisms (as is the assertion) while the hypotheses of the earlier theorems are not. In its original form for Hamiltonians on a linear symplectic space, the Weinstein conjecture was proved by Viterbo [Vi1]. Since then, the conjecture has been established for many other symplectic manifolds (sometimes under additional requirements on the level); see, e.g., [FHV, HV1, HV2, LT, Lu1, Lu2, Lu4, Vi4], to mention several results. Among these manifolds are products of complex projective spaces, manifolds of the form P × Cn (where P is compact symplectic and the product is given a split symplectic structure), and subcritical Stein manifolds. However, in general, the conjecture is still neither proved nor disproved. For example, the Weinstein conjecture in its full generality is open for cotangent bundles and T4 . Starting from the Weinstein conjecture, one can go in two different directions. One direction is to dispose of the Hamiltonian and the ambient symplectic manifold and focus exclusively on the level of contact type. This naturally leads to the question of whether a Reeb flow on a compact contact manifold necessarily has a periodic orbit; see, e.g., [Ho3]. Along these lines, Hofer [Ho2] proved the existence of periodic orbits for the Reeb flow of a contact form on S 3 or on a closed three-dimensional contact manifold M with π2 (M) = 0, and also for the Reeb flow of an overtwisted contact form. This approach interprets the conjecture as a question about the dynamics of Reeb flows and leads to the notions of contact homology and symplectic field theory [EGH, BEHWZ]. Another direction is to view the conjecture as a question about the dynamics of Hamiltonian flows on the ambient symplectic manifold. This is the perspective with which we are concerned here. More specifically, we focus on such problems as whether and how the assumption that the level has contact type can be relaxed, whether the existence of periodic orbits is typical, and so on. The contact type requirement cannot be dropped entirely: there exists a proper function on R2n (C ∞ -smooth if 2n ≥ 6 and C 2 -smooth if 2n = 4) with a regular level carrying no periodic orbits; see [Gi1, Gi3, GG1, GG2, He1, He2, Ke2]. (Constructions of such functions are known as counterexamples to the Hamiltonian Seifert conjecture.) Nevertheless, the existence of periodic orbits on the level sets of a fixed Hamiltonian is a generic phenomenon: almost all (in the sense of measure theory) regular levels of a C 2 -smooth proper function on R2n carry periodic orbits of the Hamiltonian

Weinstein conjecture and theorems of nearby/almost existence

141

flow. This result, due to Hofer and Zehnder and to Struwe, is known as the almost existence theorem [HZ3, St]. The almost existence theorem holds for many but not all symplectic manifolds (sometimes under some additional restrictions on the Hamiltonian; see [GG3]). For example, the theorem holds for CPn , products P × Cn with split symplectic structure (where P is geometrically bounded) [HV1, Lu1, MDSl, Schl], subcritical Stein manifolds [Ci, Ke3, Lu1], and small neighborhoods of certain non-Lagrangian submanifolds [Ke3, Sc3, Schl]. However, as has been observed by Zehnder [Ze], the almost existence theorem fails for certain Hamiltonians on T2n equipped with an irrational symplectic structure (Zehnder’s torus). In fact, for this Hamiltonian system, there is an interval of energy values without periodic orbits. Moreover, this phenomenon is stable under C k -small (k > 2n) perturbations of the Hamiltonian [He3, He4]. A sibling of the almost existence theorem is the theorem of dense or nearby existence which guarantees the existence of periodic orbits for a dense set of energy levels or, equivalently, near a fixed level; see, e.g., [CGK, FH, FS, HZ2, HZ3]. Both of these theorems imply the Weinstein conjecture and below we will discuss the relation between these theorems. Another reason to consider the almost existence and nearby existence theorems is that a broad class of Hamiltonian systems for which energy levels fail to have contact type naturally arises in classical mechanics. In this class are, for example, the systems describing the motion of a charge in a magnetic field, which we will discuss shortly; see also [Gi2]. For such systems one can expect the almost existence theorem to hold and periodic orbits to exist for all low-energy values. However, periodic orbits need not exist on all energy levels even when the symplectic form is exact near a level (the horocycle flow; see Example 4.7). Furthermore, as has been pointed out by Kerman [Ke1], the analysis of such systems is closely related to a generalization of the Weinstein–Moser theorem [Mo, We2]. The Weinstein–Moser theorem asserts that a smooth function H on R2n attaining a nondegenerate minimum at the origin must have at least n distinct periodic orbits on every level near the origin [Mo, We2]. Let us now replace R2n by an arbitrary symplectic manifold W and the nondegenerate minimum at one point by a Morse–Bott nondegenerate minimum along a closed symplectic submanifold M ⊂ W . Then, conjecturally, every level of H near M carries at least one periodic orbit or even a number of periodic orbits. We will refer to this conjecture as the generalized Weinstein–Moser conjecture. As a particular example motivating our interest in this question, consider π the standard kinetic energy H on the cotangent bundle W = T ∗ M → M, equipped with a twisted symplectic structure ω0 + π ∗ , where ω0 is the standard symplectic structure dp ∧ dq and is a closed two-form on M. This system describes the motion of a charge on M in the magnetic field ; see [Gi2]. When is nondegenerate M turns into a symplectic submanifold of W . The generalized Weinstein–Moser conjecture has been proved in a number of particular cases [GK1, Ke1], but in general the question is still open. Recently, however, some progress has been made along the lines of the almost existence theorem. Namely, it has been shown that almost all levels close to M of a function H attaining a minimum along M carry contractible periodic orbits [CGK, GG3, Ma2]—this is the

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relative (with respect to M) almost existence theorem for small energy values. (Note that unless M is a Morse–Bott nondegenerate minimum of H , we cannot expect such periodic orbits to exist on all levels near M [GG3].) This implies the almost existence theorem for low-energy periodic orbits of a charge in a nondegenerate magnetic field. Moreover, under suitable additional hypothesis, the genuine, nonrelative, almost existence theorem holds near M [Ke3]. In the setting of magnetic fields, these results can be further refined: periodic orbits must exist whenever = 0 [Schl]. (We will briefly discuss the proof of this result in Section 3.5.) We also refer the reader to [GK2, Ma1, Pol2] for related results. The nearby existence theorem is weaker and often easier to prove than the almost existence theorem. The pattern has been that, in many cases, the nearby existence theorem was proved first and then followed by the almost existence theorem; see, e.g., [HZ1], [HZ3, St], [CGK], and [GG3]. As we have pointed out above, both theorems imply the Weinstein conjecture. Conversely, essentially every proof of a particular case of the Weinstein conjecture in the Hamiltonian setting translates into a proof of either the nearby existence or almost existence theorem, although it is not always easy to establish which of these theorems is proved. As of today, almost existence is verified in virtually all the cases where the nearby existence has been proved. Probable exceptions are some of the results from [Vi4] on periodic orbits in cotangent bundles and, perhaps, the results of [LT] and hence of [Lu2, Lu3, Lu4]. Organization and contents of the paper In this paper we focus on the aspects of the Weinstein conjecture related to global Hamiltonian dynamics, and hence our treatment of the conjecture in general is by no means comprehensive. For example, we do not even touch upon the Weinstein conjecture for contact manifolds. (The reader interested in this conjecture is referred to the surveys [Ho3, Ho4, Ho5] in addition to the references given above.) Furthermore, we do not mention the fruitful connection between the Weinstein conjecture and Gromov–Witten invariants, although we do discuss the holomorphic curve approach to the proof of the conjecture. In Sections 2 and 3 we outline methods of proving the nearby existence and almost existence theorems and, hence, the Weinstein conjecture. These sections can be viewed as a brief introduction to certain concepts of symplectic topology (action selectors, constructions of symplectic capacities, Hofer’s metric, symplectic homology, etc.), albeit strictly focused on a specific task and not even mentioning many aspects of the subject. However, these sections should not be taken as an introduction to symplectic topology in general. For example, we assume the reader’s familiarity with Floer homology. Section 4 concerns some simple, but apparently not present in the literature, properties of the Hofer–Zehnder capacity function. Although the paper is complemented by an extensive bibliography, the list of references contains only the papers immediately relevant to our discussion. Inevitably, this list is incomplete and omits many important contributions to the subject, and our exposition emphasizes the publications that have most influenced the author’s thinking.


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Conventions In this paper, all manifolds are assumed to be without boundary.Asymplectic manifold W will be called convex if W is either closed (i.e., compact) or open and convex at infinity. Here W is said to be convex at infinity if there exists: a hypersurface ⊂ W which separates W into one set with compact closure and another, U , with noncompact closure; and a flow ϕt (for t ≥ 0) of symplectic dilations on U , which is transversal to ∂U = . Recall also that (W, ω) is symplectically aspherical if c1 |π2 (W ) = ω|π2 (W ) = 0. (In some instances, this condition can be replaced by ω|π2 (W ) = 0.) We refer the reader to, e.g., [AL, CGK] for a discussion of geometrically bounded symplectic manifolds and to [HZ3, MDSa1, MDSa2, Pol3] for a general introduction to symplectic topology. Let us now fix the sign conventions in the definition of the action functional. Let H ∈ C ∞ (S 1 × W ) and let x : S 1 → W be a contractible loop in W . Here we will use the action functional AH defined as AH (x) = − x¯ ∗ ω + H (t, x)dt, D2

S1

where x¯ : → W is a map of a disk, bounded by x. By the least action principle, contractible one-periodic orbits of H are precisely the critical points of AH . The action spectrum S(H ) of H is the set of critical values of AH , i.e., the collection of action values of AH on the contractible periodic orbits. (Since we are assuming that ω|π2 (W ) = 0, the action AH is single valued. Otherwise, one has to pass to a suitable covering of the loop space and deal with numerous other technical difficulties.) We set Ht = H (t, ·), where t ∈ S 1 , and denote by XH the Hamiltonian vector field of H . D2

2 Nearby existence theorems Nearby existence theorems are usually proved by Floer homological methods. Below we discuss some of these methods, focusing on the key ideas and omitting many (often quite nontrivial) technical details. Throughout this section, all ambient symplectic manifolds (W, ω) are assumed to be convex and symplectically aspherical, unless explicitly stated otherwise as is, for example, in Section 2.4. The argument is particularly transparent for open manifolds which are convex at infinity. Hence we consider this case first. 2.1 The action selector method: Convex at infinity open manifolds In this section we focus on convex at infinity open manifolds and outline the approach to the proof of the nearby existence theorem utilizing the notion of an action selector. In our proof of the existence of an action selector and its properties, we mainly follow [FS, Sc3]. However, many elements of our argument are already contained in [HZ2, HZ3], where the action selector is defined differently; see also, e.g., [Oh2, Vi3].

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2.1.1 Action selectors and nearby existence theorem Let W be a convex at infinity open symplectic manifold. We denote by HU , where U is an open subset of W , the space of compactly supported smooth Hamiltonians H : S 1 × U → R. For our purposes, it is convenient to adopt the following definition. An action selector is a C 0 -continuous function σ : HW → R such that1 (AS1) σ (H ) ∈ S(H ), (AS2) σ is monotone, i.e., H1 ≤ H2 implies that σ (H1 ) ≤ σ (H2 ), and (AS3) σ (H ) = max H , when H is a C 2 -small function on W with a unique maximum. Let us point out some consequences of (AS1)–(AS3) which are essential for what follows. First, recall that the action spectrum S(H ) is compact and nowhere dense; see, e.g., [HZ3, Sc3]. (This elementary, but not entirely trivial, fact can be thought of as a version of Sard’s theorem for AH ; cf. [Zv].) Furthermore, as is easy to see, S(H ) depends only on the time-one flow ϕH of H viewed as an element of the universal cover D of the group of Hamiltonian symplectomorphisms; the homotopy to identity is given by H . (In fact, when W is symplectically aspherical, S(H ) depends only on the time-one flow of H regarded as an element of the group of symplectomorphisms.) Then it follows from (AS1) and the continuity of σ that σ (H ) also depends only on ϕH ∈ D. Furthermore, σ (H ) > 0

when H is nonnegative and nonconstant,

(2.1)

by (AS2) and (AS3) and, by (AS1) and (AS2), σ (H ) = 0 when H ≤ 0. The nearby existence theorem for functions on U ⊂ W can be (and often is) easily derived from the existence of an action selector σ which meets one additional requirement that σ be a priori bounded on HU . To state the result, it is convenient to introduce the notion of a shell or thickening of a hypersurface. A shell {s } in U is an embedding × (−, ) → U , where is a closed manifold such that dim = dim U − 1. We identify × (−, ) with its image, set s = × s and assume, in addition, that = 0 divides U into two components: one bounded (i.e., such that its closure in U is compact) and the other bounded or unbounded. (In many instances, this assumption can be omitted.) The following, nearly trivial, proposition sums up a number of versions of the nearby existence theorem. Proposition 2.1. Assume that there exists an action selector σ : HW → R such that σ (K) ≤ CU for every function K ∈ HU and some constant CU independent of K. Then the nearby existence theorem holds for proper functions H on U : contractible 1 The properties (AS1)–(AS3) should not be taken as an attempt to axiomatize the notion

of an action selector (see [FGS])—such axioms would almost certainly be different from (AS1)–(AS3) and would include a version of the inequality (2.4) below. Our objective is to list the properties of the action selector that are most essential for the proof of the nearby existence theorem.


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in W periodic orbits exist for a dense set of values of H . Equivalently, for every shell {s } there exists a value s0 such that s0 carries a contractible in W closed characteristic.2 As we will soon see, there exists an action selector on R2n which is a priori bounded on bounded domains [HZ3] and hence the nearby existence theorem holds for R2n . Remark 2.2. In this proposition and in Proposition 3.1, the assumption that the shell divides W is not essential; see [MS]. Proof of Proposition 2.1. Given a shell {s }, consider a smooth function F on W such that • •

F is equal to some positive constant C > CU on the bounded component of the complement to the shell and is identically zero on the unbounded component, within the shell, F depends only on s and is a monotone decreasing function with range [0, C] and such that 0 and C are the only critical values of F .

Note that the only critical values of F on W are again 0 and C. Furthermore, 0 < σ (F ) < C by (2.1) and since σ (F ) ≤ CU < C. Hence, any contractible one-periodic orbit of F with action σ (F ) must be nontrivial and lie on one of the regular levels of F , i.e., on some hypersurface s0 . Hence, at least one of these hypersurfaces carries a contractible in W closed characteristic.

2.1.2 The existence of an action selector Let us turn now to the problem of the existence of an action selector. There are numerous constructions of action selectors for different classes of manifolds W : in [HZ2, HZ3] an action selector has been constructed for W = R2n using a direct variational method on the space of H 1/2 -loops; in [Vi3] an action selector has been defined for cotangent bundles using generating functions; this construction has been extended to Lagrangian submanifolds in [Oh1, Oh2] using Floer homology; in [Sc3, Oh2] an action selector has been introduced for symplectically aspherical closed manifolds W , again by utilizing the Floer homology methods; these results have been extended to convex at infinity manifolds in [FS]. Finally, in [Oh3], an action selector was defined for closed symplectic manifolds which are not necessarily convex or symplectically aspherical. Let us now outline the construction of an action selector, following mainly [FS, Sc3], for open symplectically aspherical manifolds that are convex at infinity. Let W be such a manifold. Recall that the Floer homology HF(H ) for H ∈ Cc∞ (S 1 ×W ) is defined and independent of H , i.e., for any two functions these groups are canonically isomorphic [Fl1, Fl2]; see also [PSS, Sa, Sc1]. Since W is not closed but convex at infinity, one has to extend H to a function with a suitable growth at 2 Depending on whether this result is thought of in terms of H or a shell, it is referred to as a

dense existence or nearby existence theorem.

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infinity, without creating new periodic orbits, and then work with the Floer homology of the resulting function; see [FS, Oh1, Vi4]. Moreover, HF(H ) is isomorphic to H∗ (W ) up to a shift of degrees, but this fact and the specific nature of the isomorphism are not very essential for us until later stages of the argument. At the moment, one may interpret H∗ (W ) as a common notation for the groups HF(H ) identified with each other for different functions H . Furthermore, the filtered Floer homology HF[a,b) (H ) is defined for any interval [a, b) with endpoints outside of S(H ). This homology is constant under deformations of a, b and H as long as a and b are outside of the action spectrum of H , see, e.g., [Vi4]. There is a natural map j a : H∗ (W ) = HF(H ) → HF[a,∞) (H ) induced by the quotient of complexes. Fix a nonzero element u ∈ H∗ (W ) and set σu (H ) = inf {a | j a u = 0}. It is easy to see by using the invariance and monotonicity properties of Floer homology that σu meets the requirements (AS1) and (AS2). Let [max] ∈ H∗ (W ) be the class of the maximum of a C 2 -small bump function. By calculating the Floer homology of such a bump function, one can show that [max] = 0. The selector σ = σ[max] obviously satisfies (AS1)–(AS3). However, the C 0 -continuity of σ , or in general of σu , requires a proof (see, e.g., [Oh2, Sc3]) and this proof relies on the explicit construction of Floer’s continuation map. The key to the proof is the following observation. Let H0 ≥ H1 be two Hamiltonians whose one-periodic orbits are nondegenerate. Consider periodic orbits x0 of H0 and x1 of H1 such that there exists a connecting homotopy trajectory joining x0 and x1 for a certain “linear’’ monotone homotopy from H0 to H1 . Then AH0 (x0 ) − AH1 (x1 ) ≤

1

max H0 (t, p) − H1 (t, p) dt.

0 p∈W

(2.2)

This inequality can be obtained by a direct calculation and the C 0 -continuity of σ readily follows from (2.2); see [Sc3] for details. In a similar vein, (2.2) implies the inequality σ (H ) ≤

1

max H (t, p)dt,

0 p∈W

(2.3)

which can be established by setting H = H0 in (2.2), taking a C 2 -small function as H1 and then letting H1 go to zero. 2.1.3 An a priori bound for σ One class of domains U for which σ is a priori bounded is the class of displaceable domains, i.e., U such that there exists a Hamiltonian symplectomorphism ϕH with


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H ∈ HW moving U away from itself: ϕH (U ) ∩ U = ∅. For example, bounded open subsets of R2n are displaceable. To show that σ is a priori bounded on a displaceable domain U , one argues as follows. t and ϕ t be time-dependent Hamiltonian flows generated by H and K in Let ϕH K t ◦ ϕ t , i.e., HW . Denote by H #K ∈ HW the Hamiltonian generating ϕH K t −1 ) (p)). H #K(t, p) = H (t, p) + K(t, (ϕH

The crucial feature of the selector σ defined in Section 2.1.2 is that σ is subadditive: σ (H #K) ≤ σ (H ) + σ (K)

(2.4)

or more generally σu∩v (H #K) ≤ σu (H ) + σv (K), where u ∩ v is the intersection of homology classes u and v. The subadditivity of σ is proved in [Oh2, Sc3] by making use of the pair-of-pants product introduced in [Sc2]; see also [PSS]. This is a product HF[a,∞) (H ) ⊗ HF[b,∞) (K) → HF[a+b,∞) (H #K) which is intersection of cycles on the full Floer homology H∗ (W ) and such that the corresponding diagram commutes. (At this stage one specifically utilizes the isomorphism HF(H ) → H∗ (W ) defined in [PSS], for this isomorphism sends the pair-of-pants product to the intersection of cycles. However, it might also be possible to prove the subadditivity of σ[max] by using the Floer continuation map.) Once the existence of such a product is established, (2.4) follows from the definition of σ ; see [Sc3, Section 4]. The subadditivity of σ implies an a priori bound for σ . Let K be a Hamiltonian whose time-one flow displaces supp H , where, by definition, supp H = , t )−1 so that supp Ht . Denote by K − the Hamiltonian generating the flow (ϕK 1 t∈S − K#K = 0. Then σ (H ) ≤ σ (K) + σ (K − ). (2.5) To prove (2.5), we argue as in [FS]. First, observe that since ϕK displaces supp H , oneperiodic orbits of H #K are exactly one-periodic orbits of K, and, as a consequence, S(H #K) = S(K). The same is, of course, true when H is replaced by the Hamiltonian sH with s ∈ R, i.e., S((sH )#K) = S(K). By continuity of σ and “discontinuity’’ of S(K), we conclude that σ ((sH )#K) ∈ S((sH )#K) = S(K) is independent of s. Setting s = 0 and s = 1 yields σ (K) = σ (H #K). Therefore, σ (H ) = σ (H #K#K − ) ≤ σ (H #K) + σ (K − ) = σ (K) + σ (K − ), which proves (2.5). Among other important examples of displaceable domains U are small neighborhoods of closed non-Lagrangian submanifolds of middle dimension whose normal bundles have nonvanishing sections [LS, Pol1]. This (combined with Macarini’s stabilization trick, [Ma1]), leads to a local version of the nearby existence theorem for twisted cotangent bundles over surfaces (other than the torus) or, in higher dimensions, for exact magnetic fields; see [FS].

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2.2 The action selector method: closed manifolds In this section we will briefly point out changes required in the action selector proof of the nearby existence theorem when W is a closed manifold. First, let us observe that the construction of an action selector outlined in Section 2.1.2 carries over to Hamiltonians on closed manifolds W. (Here, as everywhere in this section, W is assumed to be symplectically aspherical.) Such an action selector has the property σ (H + const) = σ (H ) + const and hence is never a priori bounded. To circumvent this problem, one chooses a suitable normalization of Hamiltonians. (This is also necessary to ensure that σ (H ) depends only on ϕH .) However, in contrast with open manifolds where compactly supported Hamiltonians are automatically normalized, there appears to be no natural choice of normalization for closed manifolds. One possible choice is to restrict the action selector to Hamiltonians vanishing on a neighborhood of a fixed point. This should allow one to extend word-for-word the results and constructions of Section 2.1 to closed manifolds. However, certain details of this approach are still to be worked out and we leave its discussion for a later occasion. Here, we use the traditional normalization requiring the mean value of Hamiltonians to be zero. Morespecifically, let HW be the class of smooth functions on S 1 × W normalized so that W Ht ωn = 0 and let HU be formed by Hamiltonians H ∈ HW such that supp XHt ⊂ U for all t ∈ S 1 . Proposition 2.1 still holds when the class HU is defined in such a fashion. However, when W is closed, obtaining an a priori bound for a selector on HU is more difficult than in the case of an open manifold, even though this still might be possible. We refer the reader to [FGS] for a detailed analysis of this question. (The proof of the a priori bound from Section 2.1.3 does not go through because inequality (2.5) need not hold. The reason is that even when W U is connected, S(H #K) will differ from S(K) by the constant equal to H |W U .) Here, following [Sc3], we choose a somewhat different approach. Let, as in Section 2.1.2, σ[max] be the action selector associated with the Floer homology class [max] ∈ H∗ (W ) corresponding to the maximum of a C 2 -small bump function (shifted to have zero mean). Set γ (H ) = σ[max] (H ) + σ[max] (H − ). Equivalently, γ (H ) = σ[max] (H ) − σ[min] (H ), where σ[min] is the action selector associated with the Floer homology class [min] ∈ H∗ (W ) corresponding to the minimum of a negative C 2 -small shifted bump function. Similar to action selectors for normalized functions, γ (H ) depends only on ϕH ∈ D. 1 When H is C 2 -small, we have γ (H ) = 0 (max H − min H )dt. Furthermore, γ in H , subadditive, but not necessarily monotone. Then, since is still C 0 -continuous t −1 Ht− (p) = −Ht (ϕH ) (p) , inequality (2.3) translates to γ (H ) ≤ 0

1

max H (t, p) − min H (t, p) dt. p∈W

p∈W

(2.6)


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Note also that γ (K − ) = γ (K). As we have pointed out above, the proof of (2.5) given in Section 2.1.3 does not go through for the normalization we use here. However, a similar but more involved argument proves the upper bound γ (H ) ≤ 2γ (K),

(2.7)

where the time-one flow of K displaces U ⊃ supp(XH ). (Here, by definition, , supp(XH ) = t∈S 1 supp XHt .) We refer the reader to [Sc3] for detailed proofs of these facts. Observe now that Proposition 2.1 holds when an a priori bounded selector σ is replaced by γ which satisfies (2.6) and is a priori bounded on U . (To see this, only minor modifications in the proof are needed.) As a consequence of (2.7), we immediately obtain the nearby existence theorem for displaceable domains in compact symplectically aspherical manifolds. 2.3 Limitations of the action selector method The class of manifolds W and domains U to which the action selector method applies is rather limited. For example, a bounded selector or a bounded function γ do not exist for U = W = T2 (nor for T4 or T2 ×S 2 with split symplectic structure). Indeed, it is easy to see that there is a function H ∈ HT2 with S(H ) = {min H, max H } and such that σ[max] (H ) = max H and σ[min] (H ) = max H are both arbitrarily large. The same is true for tubular neighborhoods of the zero section in cotangent bundles of some compact manifolds (e.g., of surfaces with genus g ≥ 1). As a consequence, Proposition 2.1 cannot be applied to prove nearby existence on these manifolds as long as the standard Floer homology (even accounting for noncontractible orbits) is employed. This is the case already for W = T2 even though every regular level of H is comprised of (not necessarily contractible) periodic orbits. The problem is that the periodic orbit can “migrate’’ from one homotopy class to another depending on the function in question. Another class of manifolds to which this method does not apply is formed by geometrically bounded, but not convex manifolds. Among such manifolds are many twisted cotangent bundles and also universal coverings of some manifolds, which justifies the interest in this class. The problem is that there is no known satisfactory definition of an action selector for general geometrically bounded manifolds. For example, the obstacle in the homological approach is that HF[a,b) (H ) for H ∈ HW has been defined only for intervals [a, b] which do not contain zero, while the homological definition of σ requires HF[a,b) (H ) to be defined for all intervals. One possible solution is to consider an action selector only on the class of nonnegative (autonomous or time-dependent) Hamiltonians or a yet more narrow class of functions (containing the functions F from the proof of Proposition 2.1) and to extend the homological definition to this class. The proof of the a priori bound outlined in this section will not carry over to such a narrow class, but a different argument (e.g., akin to the symplectic homology method from Section 2.4) may.

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Furthermore, when a geometrically bounded manifold is “asymptotically convex,’’ as are for instance twisted cotangent bundles, one should be able to define Floer homology for all intervals of action by suitably extending the function at infinity as in the convex case. When this is done, many of the results that hold for convex manifolds should remain valid, although certain technical difficulties have to be dealt with. However, no work in either of these directions has yet been carried out and it is not clear whether or not this would lead to new results. 2.4 Symplectic homology A slightly different approach to proving the nearby existence theorem, which also utilizes Floer homology, relies on symplectic homology introduced and investigated in [CFH, CFHW, FH, FHW]. Let, as above, U be a domain in a symplectic manifold W . The symplectic homology of U is defined as SH[a,b) (U ) = lim HF[a,b) (H ), ← − H

where the inverse limit is taken over all H ∈ Cc∞ (S 1 × U ). The symplectic homology of U detects closed characteristics in an arbitrarily narrow thickening {s } of = ∂U , provided that is smooth. In particular, when SH[a,b) (U ) = 0, in any thickening {s } there exists a hypersurface s0 carrying a closed characteristic. (This fact is an essentially immediate consequence of the definition; see [FH].) Therefore, the nearby existence theorem holds for a function H whenever the symplectic homology of the sublevels {H < c} is nontrivial. The problem is thus reduced to verifying that symplectic homology does not vanish. Let us show how this approach works, for example, when W = R2n . Let U be a bounded domain in R2n which we assume to contain the origin. Thus, there exist two open balls Br and BR centered at the origin and such that Br ⊂ U ⊂ BR . The symplectic homology has a natural monotonicity property: an inclusion U ⊂ V induces a map SH[a,b) (V ) → SH[a,b) (U ). The map # : SH[a,b) (BR ) → SH[a,b) (Br ) factors as SH[a,b) (BR ) → SH[a,b) (U ) → SH[a,b) (Br ), and hence SH[a,b) (U ) = 0 when # = 0. The symplectic homology of a ball and the map # can be calculated explicitly (see [FHW, Her1]) and, indeed, it turns out that # = 0 for some b > a > 0 and the nearby existence in R2n follows. Today, this calculation can be carried out particularly easily (see [BPS, CGK]) if one makes use of Poz´ niak’s theorem giving Floer homology in the Morse–Bott nondegenerate case [Poz]. This method also applies in the setting of the generalized Weinstein–Moser theorem discussed in the introduction. Let U be a neighborhood of a closed symplectic submanifold M of a geometrically bounded symplectically aspherical manifold W . Then, by taking suitably defined symplectic tubular neighborhoods of M as Br and


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BR , one can show that SH[a,b) (U ) = 0 [CGK]. This leads to a proof of a nearby existence theorem for narrow shells enclosing M or small values of functions having a minimum (say, equal to zero) along M. Note that since here we utilize Floer homology only for intervals that do not contain zero, the method can be used for geometrically bounded manifolds which are not necessarily convex. Furthermore, this method can also be cast in the framework of energy selectors defined on a suitable class of functions (see [Her1]). However, the benefits of this approach are unclear and we omit the details here. Remark 2.3 (stability of the area spectrum [CFHW]). As a side remark, let us mention one more application of symplectic homology and Poz´ niak’s theorem. Here, again, we focus on the main idea of the argument rather than on a complete proof. Let be a smooth hypersurface in W . The area (or action) spectrum A() is the collection of symplectic areas bounded by contractible closed characteristics on , including iterated closed characteristics. It is not hard to see using Poz´ niak’s theorem that when is the boundary of an open domain U , A() = {a ∈ R | SH[a−,a+) (U ) = 0 for any small > 0}, provided that has contact type and all (iterated) closed characteristics on are nondegenerate. (An additional, more subtle, argument is needed here when different closed characteristics bound equal areas.) Observing that the right-hand side of this equality depends solely on U , we conclude that under these hypotheses A() is determined by U . This is the stability of the area spectrum theorem [CFHW]. More specifically, let and be smooth contact type hypersurfaces in W bounding open domains U and U , respectively. Assume that all (iterated) closed characteristics on and are nondegenerate and that there exists a symplectomorphism of W sending U to U . Then A() = A( ). 2.5 Other applications In this section we briefly discuss some other applications of the action selector, which are important for what follows. 2.5.1 Homological capacity An action selector σ can be used to introduce an invariant, the homological capacity chom (U ), of a domain U in a symplectic manifold W . Assume first that W is open and convex at infinity. To an action selector σ on W , we associate a function chom on open subsets of W by setting chom (U ) = sup{σ (H ) | H ∈ HU } ∈ (0, ∞]. By definition, chom (U ) < ∞ if and only if σ is a priori bounded on U , and hence the nearby existence theorem holds for U . When W is closed, we set

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chom (U ) = sup{γ (H ) | H ∈ HU } ∈ (0, ∞]. The homological capacity is invariant under symplectomorphisms of W , monotone with respect to inclusions of domains, and homogeneous of degree one with respect to scaling of ω, i.e., chom (U, λω) = |λ| chom (U, ω) for any nonzero λ ∈ R. Here we do not touch upon the general definition and properties of symplectic capacities and refer the reader to, e.g., [Ha, Her1, Her2, Ho1, HZ2, HZ3] for a detailed discussion of this subject. In what follows we will always assume that chom is associated to σ = σ[max] or γ = σ[max] − σ[min] . Then, it is not hard to show that chom (BR ) = π R 2 by calculating the Floer homology of bump functions on BR (see [FHW] and Section 2.4). Similarly, chom (S 2 ) = area(S 2 ). However, chom (W ) = ∞, when W is a closed orientable surface other than S 2 or W = T2 × S 2 or W = T4 . In Section 3.3 we will utilize the homological capacity chom as an upper bound for the Hofer–Zehnder capacity. 2.5.2 Hofer’s geometry Denote by D the universal cover of the group of Hamiltonian symplectomorphisms of W . To be more precise, D is formed by time-one flows ϕK of Hamiltonians K ∈ HW , where each ϕK comes together with the homotopy class (with fixed end points) of t for t ∈ [0, 1]. Hofer’s norm · is defined as the path ϕK H

1

K H =

(max Kt − min Kt )dt

0

for K ∈ HW . For ψ ∈ D, set ρ(ψ) = inf { K H | K generates ψ, i.e., ψ = ϕK }. It is easy to see that ρ(ψ, ϕ) := ρ(ψϕ −1 ) is a bi-invariant metric on D, provided that ρ is nondegenerate, i.e., ρ(ψ) > 0 iff ψ = id . It turns out that ρ, known as Hofer’s metric, is indeed nondegenerate for any symplectic manifold W . Nondegeneracy of ρ has been established through a series of more and more general results starting with W = R2n (see, e.g., [HZ3]) and ending with the proof for an arbitrary W in [LMcD1]. We refer the reader to [Pol3] for an introduction to Hofer’s geometry and further references. Here we only outline the proof of nondegeneracy for symplectically aspherical convex manifolds. Assume first that W is open and convex at infinity. Let ϕK = id. Pick an open set U displaced by ϕK , i.e., such that ϕK (U ) ∩ U = ∅, and let H ∈ HU . The idea is to again utilize (2.5), but this time to obtain a lower bound for the right-hand side. Namely,


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1 1 (2.3) yields the inequality σ (K) ≤ 0 max Kt dt and also σ (K − ) ≤ − 0 min Kt dt, as can be easily seen from the definition of K − . Therefore, by (2.5), σ (H ) ≤ K H , and hence, once supp H ⊂ U and σ (H ) > 0, 0 < σ (H ) ≤ ρ(ϕK ).

(2.8)

This proves nondegeneracy of ρ for convex at infinity symplectically aspherical open manifolds. Furthermore, let us define the displacement energy of U as e(U ) = inf ρ(ψ), where ψ ∈ D displaces U . Then (2.8) translates into the upper bound chom (U ) ≤ e(U ), (2.9) which is a minor improvement over the upper bound chom (U ) ≤ 2e(U ) established in [FS]. When W is closed and symplectically aspherical, we argue in a similar fashion. Let, as above, ϕK displace U . Note that γ (K) ≤ ρ(ϕK ), by (2.6). Hence, we conclude from (2.7) that γ (H ) ≤ 2ρ(ϕK ) 1 for any H ∈ HU . When H is a C 2 -small nonzero function, γ (H ) = 0 (max Ht − min Ht )dt > 0. Therefore, ρ(ϕK ) > 0, which proves nondegeneracy of ρ. Furthermore, we also obtain the upper bound [Sc3]: chom (U ) ≤ 2e(U ).

(2.10)

In fact, the more accurate upper bound (2.9) still holds in this case; see [FGS]. Nondegeneracy of ρ for an arbitrary symplectic manifold has been established in [LMcD1] by showing, using entirely different methods, that cGr (U ) ≤ 2ρ(ϕK ), where cGr (U ) is the Gromov capacity of U , i.e., cGr (U ) = sup{π R 2 | BR symplectically embeds into U }. Note also that since cGr (U ) ≤ chom (U ), (2.8) yields that in fact cGr (U ) ≤ ρ(ϕK ), whenever W is symplectically aspherical, open, and convex at infinity.

3 Almost existence theorems Virtually all known proofs of the almost existence theorems are based on the notion of the Hofer–Zehnder capacity [HZ3], with the exception of [St] which precedes this notion.

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3.1 Hofer–Zehnder capacity and almost existence Let V be a symplectic manifold without boundary. Denote by HHZ (V ) the class of smooth nonnegative functions K on V such that • •

K is compactly supported if V is not closed or K vanishes on some open set if V is compact, K is constant near its maximum.

We will refer to such functions as Hofer–Zehnder functions. Also, let us call a nontrivial periodic orbit of K with period T ≤ 1 fast. Otherwise, an orbit will be called slow. A Hofer–Zehnder function without nontrivial fast periodic orbits will be said to be admissible. Following [HZ2, HZ3], recall that the Hofer–Zehnder capacity of V is defined as cHZ (V ) = sup{max K | K ∈ HHZ (V ) and K is admissible} ∈ (0, ∞]. The capacity cHZ (V ) does not change when the assumptions that K is nonnegative and/or that K is constant near its maximum are dropped [GG3]. The Hofer–Zehnder capacity has the same general properties as the homological capacity. One should think of cHZ as a higher dimensional analogue of the area. We will elaborate on this point in Section 4 and here we only mention that by using the area–period relation (see Section 4) one can show that for closed orientable surfaces cHZ is exactly equal to the area [Sib], in contrast with chom . The following result asserts that to prove almost existence in V , it suffices to establish that cHZ (V ) is finite. Proposition 3.1 ([HZ3]). Assume that cHZ (V ) < ∞. Then the almost existence theorem holds for proper C 2 -functions H on V : periodic orbits of H exist on almost all, in the sense of measure theory, regular levels of H . Equivalently, for every shell {s } which bounds a domain in V , the hypersurfaces s carry closed characteristics for almost all s. This proposition is a rather simple consequence of the definition of cHZ and the Arzela–Ascoli theorem; see [HZ3]. The assumption that {s } bounds a domain is superfluous [MS]. In Section 4 we will prove a more precise version of Proposition 3.1. One can also incorporate the homotopy class of an orbit in the almost existence theorem and in the definition of cHZ [Sc3]. The simplest way to do this is as follows. Fix an ambient symplectic manifold W . Let us now modify the definition of the Hofer–Zehnder capacity by requiring V to be an open subset of W and requiring K ∈ HHZ (V ) to have no nontrivial contractible in W fast periodic orbits. We denote the resulting capacity by coHZ (V ). Then Proposition 3.1 holds for contractible in W periodic orbits provided that coHZ (V ) < ∞. Clearly, cHZ (V ) = coHZ (V ), when W is simply connected, and cHZ (V ) ≤ coHZ (V ) (3.1) in general. The strict inequality is possible: for example, cHZ (S 1 ×(0, 1)) = area(S 1 × (0, 1)) < coHZ (S 1 × (0, 1)) = ∞, where we view the annulus S 1 × (0, 1) as a subset


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of itself. This also shows that the choice of the ambient manifold, even though it is not included in the notation, affects the value of coHZ . (Replace W = S 1 × (0, 1) by W = R2 .) In this connection, we also note that cHZ (U ) < ∞ for any bounded open subset U of T ∗ Tn [Ji], while coHZ (U ) = ∞ when U contains the zero section. Indeed, U can be symplectically embedded into a bounded subset of R2n since Tn admits a Lagrangian embedding in R2n . In particular, the almost existence theorem holds in T ∗ Tn . Beyond dimension two, little is known about the capacity cHZ in contrast with the capacity coHZ . For example, all results discussed in what follows deal with contractible periodic orbits and thus concern the capacity coHZ . Of course, by (3.1), an upper bound for coHZ implies an upper bound for cHZ . 3.2 Finiteness of the Hofer–Zehnder capacity In view of Proposition 3.1, to prove the almost existence theorem in V it suffices to show that cHZ (V ) < ∞. Let us start by proving that the Hofer–Zehnder capacity of a bounded domain in R2n is finite. Theorem 3.2 ([HZ2, HZ3]). Let U be a bounded domain in R2n . Then cHZ (U ) < ∞. Moreover, cHZ (BR ) = π R 2 , where BR is the ball of radius R. Proof. By monotonicity, the first assertion is an immediate consequence of the inequality cHZ (BR ) < ∞. To show that cHZ (BR ) = π R 2 , it suffices to prove that cHZ (BR ) ≤ π R 2 ; the opposite inequality is easy. (It is usually the case that establishing an upper bound for the capacity is hard while a lower bound can be easily obtained by definition.) The key is the following result. Proposition 3.3 ([HZ3]). Let H be a Hofer–Zehnder function on BR such that max H > πR 2 . Then the Hamiltonian flow of H has a nontrivial one-periodic orbit. Following [GG3], let us outline a proof of the proposition which relies on the calculation of the Floer homology and generalizes to some other situations. Let H be as in Proposition 3.3. There exist nonnegative functions K − ≤ H ≤ K + , supported in BR and depending only on the distance to the origin, and such that the action of K ± on the nearest to the origin nontrivial one-periodic orbits is greater than max K + . (These orbits are Hopf circles on a sphere enclosing the origin.) To find such functions, we make use of the assumption that H is constant near its maximum and take, as K ± , functions that squeeze H from above and below as tightly as possible and that depend only on the distance to the origin. Now, applying Poz´ niak’s theorem [Poz], one can show that HF[a,∞) (K ± ) = Z2 m for some m and a > max K + ≥ max H . This homology group is “generated’’ by the nontrivial one-periodic orbits closest to the origin. Moreover, by examining the natural homotopy from K + to K − , one can prove that the monotonicity map, which factors as

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Z2 = HF[a,∞) (K + ) → HF[a,∞) (H ) → HF[a,∞) (K − ) = Z2 , m m m [a,∞)

is an isomorphism. Hence, HFm (H ) = 0. Every trivial periodic orbit of H has action in the interval [0, max H ]. Thus, since a > max H , the flow of H must have a nontrivial one-periodic orbit. This concludes the proof of Proposition 3.3 and Theorem 3.2.

Observe that Proposition 3.3 is stronger than what is needed: the proposition guarantees the existence of a nontrivial orbit with period T = 1 while T ≤ 1 is sufficient to prove Theorem 3.2. Yet, this fact, somewhat surprisingly, appears to have no interesting applications. Also note that there are compact aspherical symplectic manifolds with infinite Hofer–Zehnder capacity. The basic example of such a manifold is Zehnder’s torus [Ze], i.e., a torus T2n with an irrational symplectic structure. All other examples of such manifolds known to the author are derivatives of Zehnder’s torus. As has been pointed out in the introduction, the nearby/almost existence theorem also fails for Zehnder’s torus. Let us now elaborate on some general principles concerning the almost existence or nearby existence theorem and the Weinstein conjecture. The existence problem for periodic orbits on a given energy level is dual in a certain, rather vague, sense to the existence problem for periodic orbits of a fixed period. The orbits of a fixed period are known to exist (Arnold’s conjecture) and a variety of methods (e.g., Floer homology) of proving this fact have been developed during the last two decades. By contrast, unless the function is assumed to be convex (and then the duality acquires a precise meaning), the problem for a fixed energy level may fail to have a solution, as counterexamples to the Hamiltonian Seifert conjecture show. Moreover, there seems to be no direct method to tackle the problem of existence of periodic orbits for a sufficiently large set of energy values (e.g., dense or full measure). All known methods, including those outlined above, first reduce the problem to proving that the flow of a function H with sufficiently large variation max H − min H possesses (nontrivial, fast, or period one) periodic orbits. Thus, all proofs of these theorems hinge on a general principle that a compactly supported function with sufficiently large variation must have fast nontrivial periodic orbits or even one-periodic orbits if the function is constant near its maximum. This principle, which is often true but fails in general (Zehnder’s torus!), can already be proved for some manifolds by utilizing, for example, Floer homology. Coming back to the discussion of the Hofer–Zehnder capacity, let us mention just one more of its properties. Namely, cHZ (ZR ) = π R 2 , where ZR = DR2 ×R2n−2 ⊂ R2n is a symplectic cylinder [HZ2, HZ3]. (Thus, the Hofer–Zehnder capacity of ZR is finite even though its volume is infinite.) This can be easily proved as follows [GG3]. First note that our proof of Proposition 3.3 readily extends to ellipsoids and shows that the capacity of an ellipsoid is equal to its minimal cross-section area (by a plane through the origin). Then exhausting ZR by more and more elongated ellipsoids we see that cHZ (ZR ) = π R 2 . The next application of our method concerns the generalized Weinstein–Moser conjecture, the motion of a charge in a magnetic field, and the relative almost exis-


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tence theorem. Let U be a neighborhood of a closed symplectic submanifold M of a geometrically bounded symplectically aspherical manifold W . Then, we can emulate the proof of Proposition 3.3 by taking, as K ± , functions that depend only on the distance to M in a suitable metric and that are supported near M. As a consequence, we obtain the relative almost existence theorem: near M, almost all levels of a function H attaining a minimum along M carry contractible periodic orbits [GG3]. (Note that this, in turn, requires replacing the ordinary Hofer–Zehnder capacity in Theorem 3.2 by its relative counterpart. The relative Hofer–Zehnder capacity cHZ (W, M), where M ⊂ W is a compact subset, is defined just as the ordinary capacity, but the function K is required to attain its maximum along M, see, e.g., [GG3, HZ2, La] for more details.) Furthermore, a more refined version of the Floer homology calculation outlined here can be used to show that coHZ (U ) < ∞ when U is a small neighborhood of a closed symplectic submanifold M with homologically trivial normal bundle in a closed symplectically aspherical manifold [Ke3]. This implies the almost existence theorem in U . o with c 3.3 Comparison of cHZ hom

In this section we will outline a different approach to obtaining an upper bound for cHZ . To be more specific, we prove that coHZ (U ) ≤ chom (U ). In our proof of this inequality we draw heavily on [HZ3, FS, Sc3], but some details appear to be new. Let W be an open manifold (with ω|π2 (W ) = 0) on which a continuous selector σ satisfying (AS1) and (AS2) is defined. Assume also that σ (H ) = max H

when H is C 2 -small and independent of time.

(3.2)

This requirement strengthens (AS3) and holds for the energy selector defined in Section 2.1.2 because the Floer complex of a C 2 -small autonomous Hamiltonian is equal to its Morse complex; see [FHS]. Let chom be the associated homological capacity. Proposition 3.4 ([FS, Sc3]). coHZ (U ) ≤ chom (U ) for any U ⊂ W . This, by (3.1), implies that cHZ (U ) ≤ chom (U ). Proof. The proposition is an immediate consequence of the following. Lemma 3.5. Let H ∈ HW be an autonomous Hamiltonian whose flow has no fast nontrivial contractible periodic orbits. Then σ (H ) = max H . To derive the proposition from the lemma, we just use the definition of the capacities: chom (U ) = sup{σ (H ) | H ∈ HU } ≥ sup{max H | H as in the lemma} = coHZ (U ).

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The assertion of the lemma is very plausible. When W is convex at infinity and σ = σ[max] , one can argue as follows. By continuity, it suffices to prove the lemma for a generic H . Then, since H does not have nontrivial contractible periodic orbits, the Floer complex of H is generated by the critical points of H and hence σ (H ) is a critical value of H . (Moreover, without loss of generality we may assume that the eigenvalues of d 2 H at the critical points of H are small. Indeed, this can be achieved by replacing H by f ◦ H , where f : R → R is a suitable diffeomorphism which is C 0 -close to identity, see [GG3, Schl]. Then σ (H ) must be the value of H at one of its local maxima, for maxima are the only critical points of H with correct index. Hence, max H = σ (H ) if H has a unique maximum.) However, to show that σ (H ) is delivered by the global maximum, one has to analyze the Floer differential of H and this indeed can be done; see, e.g., [FS, Sc3]. At this point one considers the homotopy λH with λ ∈ (0, 1] and fully uses the assumptions on H . Note also that it seems to be unknown whether in the hypotheses of the lemma fast orbits can be replaced by one-periodic orbits. One can also prove the lemma in a formal set-theoretic way, using only the continuity of σ , (AS1), (AS2) and (3.2). Denote by S the action spectrum S(H ). Observe that by the hypothesis of the lemma, every contractible one-periodic orbit of λH is trivial for all λ ∈ (0, 1], and hence the action spectrum S(λH ) is again comprised entirely of the critical values of λH . Therefore, S(λH ) = λS. Set σ (λ) = σ (λH ) ∈ λS. Then σ (λ)/λ is a continuous function of λ with values in S. Since the action spectrum S is a nowhere dense, σ (λ)/λ = const. For a small λ > 0, the function λH is C 2 small and hence σ (λH ) = max(λH ) = λ max H . It follows that σ (λ) = λ max H for all λ ∈ (0, 1] which concludes the proof of the lemma and proposition.

Proposition 3.4 also holds (see [Sc3]) when W is closed and symplectically aspherical and chom is the homological capacity defined in Section 2.5.1 for γ = σ[max] − σ[min] . This can be proved essentially in the same way as the result for open manifolds. Combining Proposition 3.4 with (2.9) and (2.10), we infer that a displaceable open set has a finite Hofer–Zehnder capacity: coHZ (U ) ≤ e(U )

if W is open,

cHZ (U ) ≤ 2e(U ) if W is closed, o

(3.3) (3.4)

whenever W is convex and symplectically aspherical. These are versions of the socalled “capacity–displacement energy inequality.’’ In particular, the almost existence theorem holds for displaceable sets. For example, let L ⊂ W be a closed nonLagrangian submanifold of middle dimension whose normal bundle has a nonvanishing section. Assume also that on W there exists a selector σ satisfying (3.2). Then, by [LS, Pol1], a small neighborhood U of L is displaceable and hence cHZ (U ) < ∞. As in Section 2.1.3, this leads to a local version of the almost existence theorem for twisted cotangent bundles over surfaces (other than the torus) or, in higher dimensions, for exact magnetic fields; see [FS, Ma1].


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Proposition 3.4 explains why the almost existence theorem can often be proved in the same setting as that of the weaker nearby existence theorem. Indeed, most of the proofs of the former, with some notable exceptions, rely on first establishing that a version of the homological capacity is finite. However, in this case the Hofer–Zehnder capacity is also finite, which implies the almost existence theorem. Remark 3.6. Proposition 3.3 suggests that in the definition of the Hofer–Zehnder capacity one may replace the condition that K has no fast periodic orbits by a weaker requirement that it has no one-periodic orbits (see [Ke3]). The resulting invariant is still a capacity. For this capacity the upper bound from Proposition 3.4 may fail to hold, unless an additional requirement on the critical set of K is imposed; see [FGS]. However, this capacity is a priori bounded on R2n and sufficient for the proof of the almost existence theorem. Furthermore, the inequality T ≤ D cH (h) in Proposition 4.2 is then replaced by the equality. (In fact, when cHZ is modified in this way, for every converging sequence cH (h) − cH (hi ) /(h − hi ) → A there exists an A-periodic orbit (not necessarily simple) on the level H = h.) As a consequence, this capacity is represented on hypersurfaces of restricted contact type in R2n (see Proposition 4.4). 3.4 Holomorphic curves and almost existence The holomorphic curve approach to the nearby existence and almost existence theorems goes back to [FHV, HV2]. Here we outline only the main idea of the method, following essentially [HV2] and omitting technical details which are in some instances quite involved. Let (W, ω) be a closed symplectic manifold and let L− and L+ be two disjoint closed submanifolds of W . Fix a generic almost complex structure J compatible with the symplectic structure and consider the space of J -holomorphic spheres u : S 2 → W in a given free homotopy class A ∈ [S 2 , W ] and with the north pole on L+ and the south pole on L− . The resulting metric space of J -holomorphic curves is not compact: the noncompact group of conformal transformations of S 2 fixing the poles acts properly on it. To make this space compact, we require that u∗ ω = ω, A /2, (3.5) D−

where D− is the southern hemisphere in S 2 . This condition eliminates the conformal flow from one pole to another, parametrized by R, and forces the resulting space M0 to be compact. This space depends on L± , A, and J . For a generic J , the space M0 is a smooth manifold and its free S 1 -equivariant cobordism class [M0 ] is independent of J . (Here the action of S 1 on M0 arises from the S 1 -action on S 2 by rotations about the vertical axis.) Note that in reality the manifold W and the class A must satisfy some additional conditions, e.g., A must be minimal, i.e., ω, A = m(W, ω); the definition of m(W, ω) is recalled below. Now let H be a smooth nonnegative function on W such that H ≡ 0 near L− and H ≡ max H near L+ . Consider the perturbed Cauchy–Riemann equation for the maps u : S 2 → W :

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∂¯J u + λ∇H = 0,

(3.6)

where λ ≥ 0 is a real parameter. Note that since ∇H = 0 in some neighborhoods of L± , this equation simply means that u is holomorphic near the poles. To make sense of this equation away from the poles, we view S 2 as the cylinder S 1 × R with the two poles attached. Then the coordinates on the cylinder are used to define ∂¯J u as a vector field along u. Let Mλ be the space of solutions of (3.6) which are in the class A, send the north and south poles to L± , and satisfy (3.5). When λ = 0, we obtain the space M0 introduced above. In general, the solutions of (3.6) can be thought of as gradient trajectories for AλH connecting trivial periodic orbits on L+ with those on L− . Then, a calculation shows that the difference of actions on these periodic orbits, which is λ max H , is bounded from above by the symplectic area of u, i.e., λ max H ≤ ω, A . As a consequence, Mλ = ∅ when λ is large. Let us examine now the disjoint union of the spaces Mλ . Under suitable genericity hypotheses, this is a smooth manifold. If this manifold is compact, it gives a cobordism from M0 to the empty set, i.e., [M0 ] = 0. Just as in Floer’s theory, compactness can fail only when a family of solutions uλ ∈ Mλ converges as λ → λ0 ≤ ω, A / max H to a broken solution which “hangs up’’ on a contractible one-periodic orbit of λ0 H , i.e., a contractible 1/λ0 -periodic orbit of H . We conclude that H must have contractible one-periodic orbits, provided that max H > ω, A and [M0 ] = 0. (Note that at this point one still has to show that the orbits found are nontrivial.) This approach leads to a few versions of the almost existence theorem, all relying on the same basic requirement that the space M0 is not cobordant to zero. In other words, the space of holomorphic curves “connecting’’ L+ and L− should be sufficiently large for the method to apply. In particular, it may be helpful to start with larger submanifolds L± or with a function H such that H ≡ 0 and H ≡ max H on large subsets. (The tradeoff is that this may result in the almost existence theorem for a restricted class of functions H .) Let us illustrate these considerations by some examples. When L± are points and the method is applicable to W and A, we conclude that cHZ (W ) ≤ ω, A and hence prove the almost existence theorem in W . There are, however, rather few manifolds W for which [M0 ] = 0 when L± are points. One example is CPn with the standard symplectic form normalized as the reduction of the unit sphere in Cn+1 . In this case the standard J is already generic, M0 = S 1 with S 1 acting by translations, and we see that cHZ (CPn ) = π [HV2]. It is also possible that this reasoning can be utilized to show that other coadjoint orbits of compact semisimple Lie groups have finite Hofer–Zehnder capacity. Now let W = P ×S 2 , where (P , β) is a compact symplectic manifold, as in [HV2]. Then taking the class of the fiber S 2 as A and applying, with some modifications, this method to L− = P × {0} and L+ = P × {∞}, one can show that the relative capacity


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cHZ (P × DR2 , P × {0}) = π R 2 as long as area(DR2 ) = π R 2 < m(P , β, J ), where u∗ β > 0 | u is a nonconstant J -holomorphic sphere . m(P , β, J ) := inf S2

In particular, m(P , β, J ) = ∞ when π2 (P ) = 0 [FHV]. Note also that m(P , β, J ) is always positive by Gromov’s compactness theorem. Furthermore, assume that ∗ 2 u β > 0 | u : S → P ≥ 0. m(P , β) := inf S2

In contrast with m(P , β, J ) ≥ m(P , β), this constant can be zero. (For instance, this is the case for P = S 2 × S 2 where the area of the first component is 1 and the second component has an irrational area.) By taking a point in P × {0} as L− and L+ as before, one can show that cHZ (P ×S 2 , L+ ) = area(S 2 ) as long as area(S 2 ) < m(P , β) [HV2]. As a consequence, cHZ (P × DR2 ) = π R 2 if π R 2 < m(P , β). (In fact, there are strong indications that cHZ (P × DR2 ) = π R 2 for any geometrically bounded symplectic manifold P and any R > 0; see [MDSl, Schl].) Symplectic manifolds P for which m(P , β) > 0 are called rational. The method also extends to the setting where P is not closed but is geometrically bounded [Lu1]. (These results have further applications to the existence problem for periodic orbits of a charge in a magnetic field, see [Ma1, Ma2].) For some other incarnations and applications of the holomorphic curve method, we refer the reader to [GL, Ke3, LT, Lu2, Lu3, Lu4]. In particular, for uniruled symplectic manifolds (such as T2 × S 2 ) and symplectic toric manifolds the Weinstein conjecture was established in [Lu2, Lu4]. In the context of the generalized Weinstein–Moser conjecture, it was proved in [Ke3] that a small neighborhood of a rational symplectic submanifold M ⊂ W has finite Hofer–Zehnder capacity coHZ . Finally, one may replace holomorphic spheres by holomorphic curves of higher genus to obtain a sufficiently large space M0 as in [LT, Lu3]. Extra care in interpreting (3.6) is then needed. For instance, imposing some additional conditions on H may be necessary, e.g., requiring H to be locally constant outside of a shell separating L− from L+ . This, depending on the details of the approach, leads to a version of either the nearby existence or almost existence theorem; see [LT, Lu2, Lu3, Lu4]. The holomorphic curve approach in the form outlined above does not apply to compact manifolds that generically have too few holomorphic curves. Among such manifolds is, for example, T4 with the standard symplectic structure. It is not known whether or not the Hofer–Zehnder capacity of T4 is finite. 3.5 Hofer’s geometry and almost existence Applications of Hofer’s geometry to nearby and almost existence theorems are based on a principle relating fast periodic orbits to minimazing properties of geodesics in t which is a one-parameter Hofer’s metric. Namely, consider the Hamiltonian flow ϕH subgroup in D and hence can be viewed as a geodesic in D. Then, conjecturally, t is length minimizing for t ∈ [0, 1), provided that H has no fast periodic orbits; ϕH

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see [MDSl] and references therein. Various particular cases of this conjecture have been proved. We refer the reader to [Pol3] for a detailed discussion and additional references and to [MDSl], following [LMcD2], for more recent results relevant to our discussion. The application of Hofer’s geometry to the circle of questions considered in this paper was pioneered in [Pol2]. Below we will just briefly indicate the logic of the argument following closely the most recent work [Schl] and in fact suppressing the connection with minimizing properties of geodesics in Hofer’s metric. Let W be a geometrically bounded symplectic manifold, which we do not require to be symplectically aspherical or convex, and let H be an autonomous Hamiltonian supported in U ⊂ W . The cornerstone of the method is the inequality coHZ (U ) ≤ 4e(U ),

(3.7)

which implies almost existence in U , provided that e(U ) < ∞. (Note that stronger inequalities (3.3) and (3.4) hold when W is symplectically aspherical and convex. Hence, the emphasis here is on extending the class of manifolds for which a version of the capacity–displacement energy inequality is proved.) The proof of (3.7) is based on the following two results: (i) Assume that supp H ⊂ U ⊂ W and H H > 4e(U ). Then ρ(ϕH ) 0. The proposition shows, in particular, that the Hofer–Zehnder capacity is strictly increasing. More specifically, we have Corollary 4.3. (i) The capacity function cH is strictly increasing. (ii) Let U and V be open bounded subsets of R2n such that U ⊂ V . Then cHZ (U ) < cHZ (V ). It is easy to see that the assumption that the sets are bounded is essential and the requirement U ⊂ V cannot be replaced by U V . Proof of Proposition 4.2. The proof of the proposition is a modification of an argument from [HZ3]. Let hi → h be a sequence such that Ai :=

cH (hi ) − cH (h) → A, hi − h


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where 0 ≤ A < ∞. By passing if necessary to a subsequence, we may assume that hi converges to h either from the right or left. In what follows we will assume that hi > h. The other case can be handled in a similar fashion. Observe that either Ai > 0 for all (sufficiently large) indexes i or cH is constant on some interval [h, h + δ], with δ > 0, since cH is monotone. Assume first that Ai > 0 and pick a sequence bi > 1 converging to one and a sequence 0 < i < (bi − 1)(hi − h)Ai . By the definition of the Hofer–Zehnder capacity, on the domain {H < h} there exists an admissible function Ki without fast nontrivial periodic orbits and such that max Ki = cH (h)−i . Let fi be a monotone decreasing function on the interval [h, hi ] identically equal to bi (hi − h)Ai near h and zero near hi and such that |fi | ≤ ai bi Ai for some sequence ai → 1+. Set Fi = fi ◦ H on the shell h ≤ H ≤ hi and smoothly extend this function to R2n by requiring it to be constant inside and outside of the shell. Then max(Ki + Fi ) = cH (hi ) + [(bi − 1)(hi − h)Ai − i ] > cH (hi ). Hence, Ki + Fi must have a nontrivial fast periodic orbit which can only be a periodic orbit of Fi . Therefore, H has a periodic orbit with period less than or equal to ai bi Ai in the shell h ≤ H ≤ hi . By passing to the limit and applying the Arzela–Ascoli theorem, we conclude that H has a periodic orbit of period less than or equal to A = lim ai bi Ai on the level H = h. To finish the proof it suffices to show that cH cannot be constant on any interval [h, h+δ]. (This will also be a direct proof of the corollary.) Assume the contrary. Then cH (hi ) = cH (h) for all large enough i. In this case we again choose a sequence of decreasing functions fi on [h, hi ] such that fi is zero near hi and a positive constant near h. (Thus fi is equal to max fi > 0 near h.) Furthermore, we can make the slope of fi so small that the function Fi has no fast nontrivial periodic orbits. Let 0 < i < max fi and let Ki be as above. It is clear that the function Ki + Fi has no fast nontrivial periodic orbits. On the other hand, we have max(Ki + Fi ) = cH (h) − i + max fi > cH (h) = cH (hi ), and hence Ki + Fi must have fast nontrivial periodic orbits. This contradiction completes the proof.

A question closely related to the area–period relation is that of representability of a capacity. Let U be the domain bounded by a compact smooth hypersurface in R2n . We say that a capacity c is represented on if there is a closed characteristic on that bounds a disc of symplectic area c(U ). For example, as is easy to see from the definition, chom is represented on smooth hypersurfaces of contact type. Since there are hypersurfaces without closed characteristics, no capacity is represented on every hypersurface. The Hofer–Zehnder capacity is represented on convex hypersurfaces [HZ2]. In fact, when is convex, cHZ (U ) is the minimal symplectic area of a closed characteristic on [HZ2]. However, it is not known if cHZ is represented on every

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contact type, or even restricted contact type, hypersurface. Arguing as in the proof of Proposition 4.2 and utilizing Lemma 3.5, one can prove the following. Proposition 4.4. Let U be the domain bounded by a smooth hypersurface of restricted contact type. Then, cHZ is subrepresented on , i.e., there exists a closed characteristic on with area less than or equal to cHZ (U ). Recall in this connection that even when U is star-shaped there can be a closed characteristic on with area strictly less than cHZ (U ); the “Bordeaux bottle’’ (see [HZ3, p. 99]) is an example. We refer the reader to, e.g., [FS, Her2] for other representability results. 4.3 Period growth and the Hofer–Zehnder capacity function As is immediately clear from the definition, the Hofer–Zehnder capacity function is necessarily continuous from the left. Beyond this trivial observation, little is known about continuity or differentiability properties of the capacity function. For example, it is not known if this function can be discontinuous at regular values. One, admittedly very naive, approach to this question is based on the estimates of the period growth. To make this more precise, fix a regular level of H , say H = 0. Let τ (h) be the infimum of all periods of periodic orbits in the open shell 0 < H < h or h < H < 0, depending on whether h is positive or negative. Then the growth of the function τ (h) is related to continuity and smoothness of cH at zero as the next proposition shows. Proposition 4.5. (i) τ (h) = O(1/ h) as h → 0+ and τ (h) = o(1/|h|) as h → 0−. (ii) Assume that τ (hk ) ≥ C/ hk for some sequence hk → 0+. Then cH (0+) − cH (0) ≥ C. (iii) Assume that τ (hk ) ≥ C/|hk |α for some sequence hk → 0 and 0 ≤ α ≤ 1. Then | cH (h) − cH (0)| ≥ C|h|1−α . The proofs of these facts follow the same line as the proof of the almost existence theorem in [HZ3]; see the proof of Proposition 4.2. Omitting a detailed argument here, we only mention that (i) is a consequence of the fact that the capacity is bounded. In fact, cHZ ({H < 0}) = ∞ if (i) fails for the left limit and cHZ (V ) = ∞ for any open set V ⊃ {H ≤ 0} if (i) fails for the right limit. Remark 4.6. The analogues of (ii) and (iii) hold when the difference of capacities is replaced by the relative capacity. Proposition 4.5 is difficult to apply to examine discontinuity or nonsmoothness of the capacity function. Indeed, let, for example, H be a Hamiltonian on R2n constructed in [Gi1, Gi3, GG1, GG2, He1, He2, Ke2] such that H = 0 carries no periodic orbits. Then cH is not Lipschitz at zero as is clear already from the results of [HZ3]. To utilize Proposition 4.5, we would need to bound from below minimal periods on the nearby levels H = h. However, the constructions of H afford little insight into the


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dynamics on these levels and obtaining such lower bounds appears to be an extremely difficult problem. Preliminary estimates indicate that cH can probably be Hölder with any α ∈ (0, 1) at H = 0 or even fail to be Hölder. However, there is no convincing evidence that cH can be discontinuous. (Note in this connection that the property of cH to be Hölder with a specific α or to be continuous, just as to be Lipschitz (see [HZ3]), is determined by the level H = 0 and is independent of the choice of H .) Consider, however, the following example. Example 4.7 (the horocycle flow). Let M be a closed surface equipped with a metric of constant negative curvature −1 and let be the area form on M. Consider the twisted symplectic structure ω = ω0 + π ∗ on W = T ∗ M, where π is the natural projection T ∗ M → M and ω0 is the standard symplectic structure. Set H = p 2 −1. The Hamiltonian flow on the level H = 0 is the horocycle flow and hence has no periodic orbits; see, e.g., [Gi2, Gi4] for details. Assume that the Hofer–Zehnder capacity of the sets {H < h} for h near zero is finite. (This is not known, although is likely to be true, even for h < 0 close to zero. For small neighborhoods of the zero section (i.e., h ≈ −1), finiteness has been recently proved in [FS]; however, for h > 0, finiteness of cHZ appears to be beyond reach of the methods considered in this paper.) Then we claim that √ cH (h) − cH (0) ≥ lmin h for h > 0, (4.1) where lmin is the minimal length of a closed geodesic on M. Therefore, cH is not smoother at h = 0 than 1/2-Hölder on the right. To prove this, let us first note that √ τ (h) = lmin / h for h > 0, (4.2) √ and hence, by (iii), cH (h) − cH (0) ≥ lmin h. Establishing (4.2) directly appears to be rather difficult. Instead, let us observe that there exists a symplectomorphism (T ∗ M {H ≤ 0}, ω) → (T ∗ M M, ω0 ) which sends p 2 to p 2 −1. (Such a symplectomorphism can be constructed, for instance, by judiciously applying Moser’s method.) This allows one to translate the period growth on (T ∗ M, ω0 ) as p → 0, which is lmin / p for the Hamiltonian p 2 /2, to the period growth on (T ∗ M, ω) for H > 0. Note also that by applying the results of [BPS] and using√the above symplectomorphism, one can prove that cHZ ({H < h}, {H ≤ 0}) ≤ lmin h. This, together with the analogue of (4.1) for the relative capacity, proves that cHZ ({H < h}, {H ≤ 0}) = √ lmin h. One can also estimate the period growth on the left. All orbits on the level H = h < 0 are closed and project to geodesic circles on M with √ geodesic curvature kg > 1. A straightforward calculation shows that τ (h) = 2π/ |h| for h < 0 and hence, by √ (iii), cH (0) − cH (h) ≥ 2π |h|. Thus, on the left, cH is again not smoother than 1/2-Hölder. Acknowledgments The author is deeply grateful to Paul Biran, Urs Frauenfelder, Ba¸sak Gürel, Ely Kerman, Debra Lewis, Leonid Polterovich, Felix Schlenk, and the referees for their useful remarks and suggestions.

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References [AL]

M. Audin and J. Lafontaine, eds., Holomorphic Curves in Symplectic Geometry, Progress in Mathematics, Vol. 117, Birkhäuser, Basel, 1994. [Ar] V. I. Arnold, Mathematical Methods of Classical Mechanics, Springer-Verlag, Berlin, New York, Heidelberg, 1984. [BPS] P. Biran, L. Polterovich, and D. Salamon, Propagation in Hamiltonian dynamics and relative symplectic homology, Duke Math. J., 119-1 (2003), 65–118. [BEHWZ] F. Bourgeois, Y. Eliashberg, H. Hofer, K. Wysocki, and E. Zehnder, Compactness results in symplectic field theory, Geom. Topology, 7 (2003), 799–888. [Ci] K. Cieliebak, Subcritical Stein manifolds are split, preprint, 2002; math.DG/ 0204351. [CFH] K. Cieliebak, A. Floer, and H. Hofer, Symplectic homology II: A general construction, Math. Z., 218 (1995), 103–122. [CFHW] K. Cieliebak, A. Floer, H. Hofer, and K. Wysocki, Applications of symplectic homology II: Stability of the action spectrum, Math. Z., 223 (1996), 27–45. [CGK] K. Cieliebak, V. Ginzburg, and E. Kerman, Symplectic homology and periodic orbits near symplectic submanifolds, Comment. Math. Helv., 79-3 (2004), 554– 581. [EGH] Y. Eliashberg, A. Givental, and H. Hofer, Introduction to symplectic field theory, Geom. Functional Anal., Special Volume, Part II (2000), 560–673. [Fl1] A. Floer, Morse theory for Lagrangian intersections, J. Differential Geom., 28 (1988), 513–547. [Fl2] A. Floer, Witten’s complex and infinite dimensional Morse theory, J. Differential Geom., 30 (1989), 202–221. [FH] A. Floer and H. Hofer, Symplectic homology I: Open sets in Cn , Math. Z., 215 (1994), 37–88. [FHS] A. Floer, H. Hofer, and D. Salamon, Transversality in elliptic Morse theory for the symplectic action, Duke Math. J., 80 (1995), 251–292. [FHV] A. Floer, H. Hofer, and C. Viterbo, The Weinstein conjecture in P × Cl , Math. Z., 203 (1990), 469–482. [FHW] A. Floer, H. Hofer, and K. Wysocki, Applications of symplectic homology I: Math. Z., 217 (1994), 577–606. [FGS] U. Frauenfelder, V. Ginzburg, and F. Schlenk, Energy capacity inequalities via an action selector, preprint, 2004; math.DG/0402404. [FS] U. Frauenfelder and F. Schlenk, Hamiltonian dynamics on convex symplectic manifolds, preprint, 2003; math.SG/0303282. [GL] D. Gatien and F. Lalonde, Holomorphic cylinders with Lagrangian boundaries and Hamiltonian dynamics, Duke Math. J., 102 (2000), 485–511. [Gi1] V. L. Ginzburg, An embedding S 2n−1 → R2n , 2n − 1 ≥ 7, whose Hamiltonian flow has no periodic trajectories, Internat. Math. Res. Notices, 1995-2 (1995), 83–98. [Gi2] V. L. Ginzburg, On closed trajectories of a charge in a magnetic field. An application of symplectic geometry, in Contact and Symplectic Geometry (Cambridge, 1994), Publications of the Newton Institute, Vol. 8, Cambridge University Press, Cambridge, UK, 1996, 131–148. [Gi3] V. L. Ginzburg, A smooth counterexample to the Hamiltonian Seifert conjecture in R6 , Internat. Math. Res. Notices, 1997-13 (1997), 641–650.

Weinstein conjecture and theorems of nearby/almost existence [Gi4]

[Gi5]

[GG1]

[GG2] [GG3] [GK1]

[GK2] [Ha] [He1] [He2]

[He3]

[He4]

[Her1] [Her2] [Ho1]

[Ho2] [Ho3]

[Ho4]

[Ho5]

169

V. L. Ginzburg, Hamiltonian dynamical systems without periodic orbits, in Northern California Symplectic Geometry Seminar, AMS Translations (Series 2), Vol. 196, American Mathematical Society, Providence, RI, 1999, 35–48. V. L. Ginzburg, The Hamiltonian Seifert conjecture: Examples and open problems, in Proceedings of the 3rd European Congress of Mathematics, Barcelona, 2000, Vol. II, Progress in Mathematics, Vol. 202, Birkhäuser, Boston, 2001, 547–555. V. L. Ginzburg and B. Z. Gürel, On the construction of a C 2 -counterexample to the Hamiltonian Seifert conjecture in R4 , Electron. Res. Announc. Amer. Math. Soc., 8 (2002), 1–10. V. L. Ginzburg and B. Z. Gürel, A C 2 -smooth counterexample to the Hamiltonian Seifert conjecture in R4 , Ann. Math., 158 (2003), 953–976. V. L. Ginzburg and B. Z. Gürel, Relative Hofer–Zehnder capacity and periodic orbits in twisted cotangent bundles, Duke Math. J., 123-1 (2004), 1–47. V. L. Ginzburg and E. Kerman, Periodic orbits in magnetic fields in dimensions greater than two, in Geometry and Topology in Dynamics (Winston-Salem, NC, 1998/San Antonio, TX, 1999), Contemporary Mathematics, Vol. 246, American Mathematical Society, Providence, RI, 1999, 113–121. V. L. Ginzburg and E. Kerman, Periodic orbits of Hamiltonian flows near symplectic extrema, Pacific J. Math., 206 (2002), 69–91. U. Hamenstaedt, Examples for nonequivalence of symplectic capacities, preprint, 2002; math.SG/0209052. M.-R. Herman, fax to Eliashberg, 1994. M.-R. Herman, Examples of compact hypersurfaces in R2p , 2p ≥ 6, with no periodic orbits, in C. Simo, ed., Hamiltonian Systems with Three or More Degrees of Freedom: Proceedings of the NATO Advanced Study Institute, S’Agaro, Spain, June 19–30, 1995, NATO Science Series C: Mathematical and Physical Sciences, Vol. 533, Kluwer Academic Publishers, Dordrecht, the Netherlands, 1999. M.-R. Herman, Examples de flots hamiltoniens dont aucune perturbations en topologie C ∞ n’a d’orbites périodiques sur ouvert de surfaces d’énergies, C. R. Acad. Sci. Paris Sér. I Math., 312 (1991), 989–994. M.-R. Herman, Différentiabilité optimale et contre-exemples à la fermeture en topologie C ∞ des orbites récurrentes de flots hamiltoniens, C. R. Acad. Sci. Paris Sér. I Math., 313 (1991), 49–51. D. Hermann, Non-equivalence of symplectic capacities for open sets with restricted contact type boundaries, preprint, Orsay, France, 1998. D. Hermann, Holomorphic curves and Hamiltonian systems in an open set with restricted contact-type boundary, Duke Math. J., 103 (2000), 335–374. H. Hofer, Symplectic capacities, in Geometry of Low-Dimensional Manifolds 2 (Durham, 1989), London Mathematical Society Lecture Notes, Vol. 151, Cambridge University Press, Cambridge, UK, 1990, 15–34. H. Hofer, Pseudoholomorphic curves in symplectizations with applications to the Weinstein conjecture in dimension three, Invent. Math., 114 (1993), 515–563. H. Hofer, Dynamics, topology, and holomorphic curves, in Proceedings of the International Congress of Mathematicians (Berlin, 1998), Extra Vol. I, Documenta Mathematica, 1998, 255–280 (electronic). H. Hofer, Holomorphic curves and dynamics in dimension three, in Symplectic Geometry and Topology (Park City, UT, 1997), IAS/Park City Mathematics Series, Vol. 7, American Mathematical Society, Providence, RI, 1999, 35–101. H. Hofer, Holomorphic curves and real three-dimensional dynamics, Geom. Functional Anal., Special Volume, Part II (2000), 674–704.

170

V. L. Ginzburg

[HV1] [HV2] [HZ1] [HZ2] [HZ3] [Ji] [Ke1] [Ke2] [Ke3] [La]

[LMcD1] [LMcD2]

[LS] [LT] [Lu1]

[Lu2] [Lu3] [Lu4] [Ma1] [Ma2] [MS] [MDSa1] [MDSa2]

H. Hofer and C. Viterbo, The Weinstein conjecture in cotangent bundles and related results, Ann. Sc. Norm. Sup. Pisa Ser. IV Fasc. III, 15 (1988), 411–445. H. Hofer, C. Viterbo, The Weinstein conjecture in the presence of holomorphic spheres, Comm. Pure Appl. Math., 45 (1992), 583–622. H. Hofer and E. Zehnder, Periodic solutions on hypersurfaces and a result by C. Viterbo, Invent. Math., 90 (1987), 1–9. H. Hofer and E. Zehnder,Anew capacity for symplectic manifolds, in P. Rabinowitz and E. Zehnder, eds., Analysis, et Cetera, Academic Press, Boston, 1990, 405–427. H. Hofer and E. Zehnder, Symplectic Invariants and Hamiltonian Dynamics, Birkhäuser Advanced Texts, Birkhäuser, Basel, 1994. M. Y. Jiang, Periodic solutions of Hamiltonian systems on hypersurfaces in a torus, Manuscripta Math., 85 (1994), 307–321. E. Kerman, Periodic orbits of Hamiltonian flows near symplectic critical submanifolds, Internat. Math. Res. Notices, 1999-17 (1999), 954–969. E. Kerman, New smooth counterexamples to the Hamiltonian Seifert conjecture, J. Symplectic Geom., 1 (2002), 253–267. E. Kerman, Semi-local symplectic topology and some global applications, in preparation. F. Lalonde, Energy and capacities in symplectic topology, in Geometric Topology (Athens, GA, 1993), AMS/IP Studies in Advanced Mathematics, Vol. 2.1, American Mathematical Society, Providence, RI, 1997, 328–374. F. Lalonde and D. McDuff, The geometry of symplectic energy, Ann. Math. (2), 141 (1995), 349–371. F. Lalonde and D. McDuff, Hofer’s L∞ -geometry: Energy and stability of Hamiltonian flows I, II: Invent. Math., 122 (1995), 1–33, 35–69; errata, Invent. Math., 123 (1996), 613. F. Laudenbach, J.-C. Sikorav, Hamiltonian disjunction and limits of Lagrangian submanifolds, Internat. Math. Res. Notices 1994-1 (1994), 161–168. G. Liu and G. Tian, Weinstein conjecture and GW invariants, Comm. Contemp. Math., 2 (2000), 405–459. G. Lu, The Weinstein conjecture on some symplectic manifolds containing the holomorphic spheres, Kyushu J. Math., 52 (1998), 331–351; addendum, Kyushu J. Math., 54 (2000), 181–182. G. Lu, The Weinstein conjecture in the uniruled manifolds, Math. Res. Lett., 7 (2000), 383–387. G. Lu, Gromov-Witten invariants and pseudo symplectic capacities, preprint, 2001; math.SG/0103195, v.6. G. Lu, Symplectic capacities of toric manifolds and related results, preprint, 2003; math.SG/0312483. L. Macarini, Hofer–Zehnder capacity and Hamiltonian circle actions, Comm. Contemp. Math., (2003). L. Macarini, Hofer–Zehnder semicapacity of cotangent bundles and symplectic submanifolds, preprint, 2003; math.SG/0303230. L. Macarini and F. Schlenk, A refinement of the Hofer-Zehnder theorem on the existence of closed trajectories near a hypersurface, Bull. London Math. Soc., (2003). D. McDuff and D. Salamon, Introduction to Symplectic Topology, Oxford University Press, New York, 1995. D. McDuff and D. Salamon, J -Holomorphic Curves and Quantum Cohomology, University Lecture Series, Vol. 6, American Mathematical Society, Providence, RI, 1994.

Weinstein conjecture and theorems of nearby/almost existence [MDSl] [Mo] [Na] [Ne] [Oh1] [Oh2] [Oh3] [Pol1]

[Pol2]

[Pol3] [Poz]

[PSS]

[Ra] [Sa]

[Schl] [Sc1] [Sc2]

[Sc3] [Sib] [Sik] [St] [Vi1]

171

D. McDuff and J. Slimowitz, Hofer–Zehnder capacity and length minimizing Hamiltonian paths, Geom. Topol., 5 (2001), 799–830 (electronic). J. Moser, Periodic orbits near equilibrium and a theorem by Alan Weinstein, Comm. Pure Appl. Math., 29 (1976), 727–747. I. P. Natanson, Theory of Functions of a Real Variable, Frederick Ungar Publishing Company, New York, 1955. E. Neduv, Prescribed minimal period problems for convex Hamiltonian systems via Hofer–Zehnder symplectic capacity, Math. Z., 236 (2001), 99–112. Y.-G. Oh, Symplectic topology as the geometry of action functional I: Relative Floer theory on the cotangent bundle, J. Differential Geom., 46 (1997), 499–577. Y.-G. Oh, Symplectic topology as the geometry of action functional II: Pants product and cohomological invariants, Comm. Anal. Geom., 7 (1999), 1–54. Y.-G. Oh, Mini-max theory, spectral invariants and geometry of the Hamiltonian diffeomorphism group, preprint, 2002; math.SG/0206092. L. Polterovich,An obstacle to non-Lagrangian intersections, in H. Hofer, C. Taubes, A. Weinstein, and E. Zehnder, eds., The Floer Memorial Volume, Progress in Mathematics, Vol. 133, Birkhäuser, Basel, 1995, 575–586. L. Polterovich, Geometry on the group of Hamiltonian diffeomorphisms, in Proceedings of the International Congress of Mathematicians (Berlin, 1998), Extra Vol. II, Documenta Mathematica, 1998, 401–410 (electronic). L. Polterovich, The Geometry of the Group of Symplectic Diffeomorphisms, Lectures in Mathematics ETH Zürich, Birkhäuser, Basel, 2001. M. Po´zniak, Floer homology, Novikov rings and clean intersections, in Northern California Symplectic Geometry Seminar, AMS Translations (Series 2), Vol. 196, American Mathematical Society, Providence, RI, 1999, 119–181. S. Piunikhin, D. Salamon, and M. Schwarz, Symplectic Floer–Donaldson theory and quantum cohomology, in Contact and Symplectic Geometry (Cambridge, 1994), Publications of the Newton Institute, Vol. 8, Cambridge University Press, Cambridge, UK, 1996, 171–201. P. Rabinowitz, Periodic solutions of a Hamiltonian system on a prescribed energy surface. J. Differential Equations, 33 (1979), 336–352. D. A. Salamon, Lectures on Floer homology, in Y. Eliashberg and L. Traynor, eds., Symplectic Geometry and Topology, IAS/Park City Mathematics Series, Vol. 7, American Mathematical Society, Providence, RI, 1999, 143–230. F. Schlenk, Applications of Hofer’s geometry to Hamiltonian dynamics, in preparation. M. Schwarz, Morse Homology, Birkhäuser, Basel, 1993. M. Schwarz, Cohomology Operations from S 1 -Cobordisms in Floer Homology, Ph.D. thesis, Dissertation ETH 11182, Swiss Federal Institute of Technology, Zurich, 1995. M. Schwarz, On the action spectrum for closed symplectically aspherical manifolds, Pacific J. Math., 193 (2000), 419–461. K. F. Siburg, Symplectic capacities in two dimensions, Manuscripta Math., 78 (1993), 149–163. J.-C. Sikorav, Systèmes hamiltoniens et topologie symplectique, ETS Editrice Pisa, Dipartamento di Matematica, Università di Pisa, Pisa, 1990. M. Struwe, Existence of periodic solutions of Hamiltonian systems on almost every energy surface, Bol. Soc. Bras. Mat., 20 (1990), 49–58. C. Viterbo, A proof of Weinstein’s conjecture in R2n , Ann. Inst. Poincaré, Anal. Non Linéaire, 4 (1987), 337–356.

172 [Vi2]

[Vi3] [Vi4] [We1] [We2] [We3] [We4] [Ze]

[Zv]

V. L. Ginzburg C. Viterbo, Capacités symplectiques et applications (d’après Ekeland–Hofer, Gromov), Astérisque, 177–178 (1989) (Séminaire Bourbaki, Vol. 1988/89), exp. 714, 345–362. C. Viterbo, Symplectic topology as the geometry of generating functions, Math. Ann., 292 (1992), 685–710. C. Viterbo, Functors and computations in Floer homology with applications I, Geom. Functional Anal., 9 (1999), 985–1033. A. Weinstein, Lagrangian submanifolds and Hamiltonian systems, Ann. Math. (2), 98 (1973), 377–410. A. Weinstein, Normal modes for non-linear Hamiltonian systems, Invent. Math., 20 (1973), 377–410. A. Weinstein, Periodic orbits for convex Hamiltonian systems, Ann. Math. (2), 108 (1978), 507–518. A. Weinstein, On the hypotheses of Rabinowitz’ periodic orbit theorems, J. Differential Equations, 33 (1979), 353–358. E. Zehnder, Remarks on periodic solutions on hypersurfaces, in P. H. Rabinowitz, A. Ambrosetti, I. Ekeland, E. J. Zehnder, eds., Periodic Solutions of Hamiltonian Systems and Related Topics, NATO Science Series C: Mathematical and Physical Sciences, Vol. 209, Reidel, Dordrecht, the Netherlands, 1987, 267–279. V. G. Zvyagin, The set of critical values of a potential Fredholm functional, Math. Notes, 63-1 (1998), 118–120.

Simple singularities and integrable hierarchies∗ Alexander B. Givental and Todor E. Milanov Department of Mathematics University of California at Berkeley Berkeley, CA 94720-3840 USA [email protected], [email protected] To Alan Weinstein on his 60th birthday. Abstract. The paper [11] gives a construction of the total descendent potential corresponding to a semisimple Frobenius manifold. In [12], it is proved that the total descendent potential corresponding to K. Saito’s Frobenius structure on the parameter space of the miniversal deformation of the An−1 -singularity satisfies the modulo-n reduction of the KP-hierarchy. In this paper, we identify the hierarchy which is satisfied by the total descendent potential of a simple singularity of ADE type. Our description of the hierarchy is parallel to the vertex operator construction of Kac–Wakimoto [17] except that we give both some general integral formulas and explicit numerical values for certain coefficients which in the Kac–Wakimoto theory are studied on a case-by-case basis and remain, generally speaking, unknown.

1 ADE-hierarchies According to Date–Jimbo–Kashiwara–Miwa [6] and I. Frenkel [10], the KdVhierarchy of integrable systems can be placed under the name A1 into the list of more general integrable hierarchies corresponding to the ADE Dynkin diagrams. These hierarchies are usually constructed (see [16]) using the representation theory of the corresponding loop groups. V. Kac and M. Wakimoto [17] describe the hierarchies even more explicitly in the form of the so-called Hirota quadratic equations expressed in terms of suitable vertex operators. One of the goals of this paper is to show how the vertex operator description of the Hirota quadratic equations (certainly the same ones, even though we don’t quite prove this) emerges from the theory of vanishing cycles associated with ADE-singularities. Let f be a weighted-homogeneous polynomial in C3 with a simple critical point at the origin. According to V. Arnold [1] simple singularities of holomorphic functions are classified by simply-laced Dynkin diagrams: ∗ This material is based on work supported by National Science Foundation grants DMS-

0072658 and DMS-0306316.

174

A. B. Givental and T. E. Milanov

x2 x2 x1N +1 + 2 + 3, N +1 2 2 N −1 2 + x32 , DN , N ≥ 4: f = x1 x2 − x2 AN , N ≥ 1: f =

E6 : f = x13 + x24 + x32 , E7 :

f = x13 + x1 x23 + x32 ,

E8 : f = x13 + x25 + x32 . Let H = C[x1 , x2 , x3 ]/(fx1 , fx2 , fx3 ) denote the local algebra of the critical point. We equip H with a nondegenerate symmetric bilinear form (·, ·) by picking a weightedhomogeneous holomorphic volume ω = dx1 ∧ dx2 ∧ dx3 and using the residue pairing ϕ(x)ψ(x)ω (ϕ, ψ) := Res0 . fx1 fx2 fx3 Let H = H ((z−1 )) be the space of Laurent series f (z) = k∈Z fk zk in one indeterminate z−1 (i.e., finite in the direction of positive k) with vector coefficients fk ∈ H . We endow H with the symplectic form . 1

(f , g) := (f (−z), g(z))dz. 2π i The polarization H = H+ ⊕ H− , where H+ = H [z] and H− = z−1 H [[z−1 ]], is Lagrangian and identifies H with the cotangent bundle space T ∗ H+ . The Hirota quadratic equations are imposed on asymptotical functions of q = q0 + q1 z + q2 z2 + · · · ∈ H+ . By an asymptotical function we mean an expression of the form = exp

∞

g−1 F (g) (q),

g=0

where usually F (g) will be formal functions on H+ . By definition, vertex operators are elements of the Heisenberg group acting on such functions. Given a sum f = fk zk (possibly infinite in both directions) one defines the corresponding vertex operator of the form √

√

e (f− ,q)/ e ∂f+ ⎫ ⎧ ⎫ ⎧ ⎬ ⎨ ⎬ ⎨√ √ a = exp (−1)k+1 f−1−k qka / exp fka ∂/∂qka . ⎭ ⎩ ⎭ ⎩ k≥0

a

k≥0 a

Here fka , qka are components of the vectors fk , qk in an orthonormal basis. We will make use of the vertex operators φ (λ) corresponding to two-dimensional homology classes φ ∈ H2 (f −1 (1)) ! ZN and defined as follows. Take

Simple singularities and integrable hierarchies

f :=

(k)

Iφ (λ)(−z)k ,

(k)

175

(k+1)

where dIφ /dλ = Iφ

k∈Z (−1)

and Iφ

(λ) ∈ H is the following period vector: (−1) (Iφ (λ), [ψa ])

1 := 2π

φ⊂f −1 (λ)

ψa (x)

ω . df

The cycle φ is transported from the level surface f −1 (1) to f −1 (λ), and ψa are weighted-homogeneous functions representing a basis in the local algebra H .1 The (k) functions (Iφ , [ψa ]) are proportional to the fractional powers λma / h−k−1 where h is the Coxeter number and ma = 1 + h deg ψa are the exponents of the appropriate reflection group AN , DN , or EN . The lattice H2 (f −1 (1)) carries the action of the monodromy group (defined via morsification of the function f ) which is the reflection group with respect to the intersection form of cycles. The form is negative definite, and we will denote ·, · the positive definite form opposite to it. Let A denote the set of vanishing cycles, i.e., the set of classes α ∈ H2 (f −1 (1)) with α, α = 2 such that the reflections φ → φ − α, φα belong to the monodromy group. The Hirota quadratic equation of the ADE type takes on the form ( ) dλ N (h + 1) α −α Resλ=∞ ( ⊗ ) (1) aα (λ) ⊗ (λ) ( ⊗ ) = λ 12h α∈A

ma ∂ ∂ + + k (qka ⊗ 1 − 1 ⊗ qka ) ⊗ 1 − 1 ⊗ ( ⊗ ). h ∂qka ∂qka a k≥0

(2) The tensor product sign means that the functions depend on two copies q and q of the variable q, and the objects on the left of ⊗ refer to q = q while those on the right to q = q . The equation can be interpreted as follows. Set q = x + y, q = x − y and expand (1), (2) as a power series in y. Namely, rewrite the vertex operators: / 0 / 0 a α (λ) ⊗ −α (λ) = exp −1/2 yka exp 2(−1)k+1 f−1−k fka 1/2 ∂yka , a where the coefficients fka (respectively, f−1−k ) are proportional to negative (respectively, positive) fractional powers of λ. The residue sum (which should be understood here as the coefficient at λ0 ) can therefore be written as a power series ym Pm (∂y ) in y with coefficients Pm which are differential polynomials. Also, ⊗ = (x + y)(x − y) can be expanded into the Taylor power series in y with coefficients which are quadratic expressions in partial derivatives of (x). Finally, the operator in (2) assumes the form 2 a,k (ma / h + k)yka ∂yka . Equating coefficients 1 As it follows, for instance, from [13], the integral on the right-hand side depends only on

the class [ψa ] ∈ H .

176


in (1), (2) at the same monomials ym , we obtain a hierarchy of quadratic relations between partial derivatives of (x). In particular, the equation corresponding to y0 shows that

aα =

α∈A

N (h + 1) 12h

(3)

is a necessary condition for consistency of the hierarchy (i.e., for existence of a nonzero solution ). According to C. Hertling (see the last chapter in [15]), for any weightedhomogeneous singularity the expressions N (h+1)/(12h) and h−2 a ma (h−ma )/2 coincide. Therefore, the operator on the right-hand side of the Hirota equation is twice the Virasoro operator2

ma (h − ma ) + k yka ∂yka + . h 4h2 a

ma a,k

The coefficients aα actually depend only on the orbit of the vanishing cycle α under the action of the classical monodromy operator defined by transporting the cycles in f −1 (λ) around λ = 0 and acting as one of the Coxeter elements in the reflection group. In fact, the root system A consists of N such orbits with h elements each. Summing the vertex operators within the same orbit acts as taking the average over all h branches of the function λ1/ h . Thus the total sum does not contain fractional powers of λ when expanded near λ = ∞. The exact values of the coefficients aα can be described as follows. To a vector β ∈ H2 (f −1 (1), C) ! CN , associate the meromorphic 1-form on CN Wβ := −

dγ , x 1 . β, γ 2 2 γ , x

(4)

γ ∈A

Let w be an element of the reflection group and α and β = wα be two roots. Then aβ /aα = exp

w−1 κ

κ

Wα =

1

κ, γ α,γ

2 /2−β,γ 2 /2

,

(5)

γ ∈A

where κ ∈ CN denotes an eigenvector of the classical monodromy operator M with the eigenvalue exp(2π i/ h). The right-hand side does not depend on the path connecting κ with w −1 κ since Wα is closed with logarithmic poles on some mirrors and with periods that are integer multiples of 2π i. It does not depend on the normalization of κ since Wα is homogeneous of degree 0. Also, the identity (see, e.g., [5, Section V.6.2]) γ , x2 = 2hx, x γ ∈A 2 In a sense it corresponds to the vector field λ∂ in the Lie algebra of vector fields on the λ

line—see Section 7 for further information about this.


177

M −h κ M −1 κ implies that i xa ∂/∂xa Wα = −2h and shows that κ Wα = h−1 κ Wα = −4π i so that aMα = aα as expected. While the ratios of aα are determined by (5), the normalization of aα is found from (3) which says that the average value of aα is (h + 1)/12h2 . Later we give two other descriptions of the coefficients aα —as certain limits and as explicit case-by-case values. Conjecture. The Hirota quadratic equation (1)–(5) coincides (up to certain rescaling of the variables qka ) with the corresponding ADE-hierarchy of Kac–Wakimoto [17]. In Section 8, we confirm this conjecture in the cases AN , D4 , and E6 .3

2 The total descendent potential The second goal of this paper is to generalize to the ADE-singularities the result of [12] that the total descendent potential associated to the An−1 -singularity in the axiomatic theory of topological gravity is a tau-function of the nKdV-hierarchy (or Gelfand–Dickey-hierarchy). According to E. Witten’s conjecture [22] proved by M. Kontsevich [18], the following generating function for intersection indices on the Deligne–Mumford spaces satisfies the equation of the KdV-hierarchy:4 ' * m ∞ 1 g−1 k ψi + (6) DA1 = exp qk ψ i . m! Mg,m g,m i=1

k=0

In the axiomatic theory, the total descendent potential is, by definition, an asymptotical function of the form D = exp g−1 F (g) (q), g≥0

where F (g) are formal functions on H+ near the point q = −1z. (Here 1 is the unit element in the local algebra H .) This convention called the dilaton shift is already explicitly present in (6). The formal functions F (g) called the genus g descendent potentials are supposed to satisfy certain axioms dictated by Gromov–Witten theory. The axioms (while not entirely known) are to include the so-called string equation (SE), dilaton equation (DE), topological recursion relations (TRR or 3g − 2-jet property), and Virasoro constraints. According to [14], the genus-0 axioms SE + DE + TRR for F (0) are equivalent to the following geometrical property (∗) of the Lagrangian submanifold L ⊂ H = T ∗ H+ defined as the graph of dF (0) : 3 There has been a new development in the subject which leads, in particular, to the proof of

the conjecture: motivated partly by this paper, E. Frenkel found a simple formula for the analogues in the Kac–Wakimoto theory of the coefficients aα . 4 Here ψ is the first Chern class of the line bundle over M g,m formed by the cotangent lines i to the curves at the ith marked points.

178


(∗) L is a Lagrangian cone with the vertex at the origin and such that tangent spaces L to L are tangent to L exactly along zL. In other words, the cone L is swept by the family τ ∈ H → zLτ of isotropic subspaces which form a variation of semiinfinite Hodge structures in the sense of S. Barannikov [3]. According to his results, this defines a Frobenius structure on the space of parameters τ . In the case of ADE-singularities (and, more generally, finite reflection groups) the Frobenius structures have been constructed by K. Saito [20]. Consider the miniversal deformation fτ (x) = f (x) + τ 1 ψ1 (x) + · · · + τ N ψN (x), where {ψa } form a weighted-homogeneous basis in the local algebra H , and ψN = 1. The tangent spaces Tτ T to the parameter space T ! CN are canonically identified with the algebras of functions on the critical schemes crit (fτ ): ∂τ a → ∂fτ /∂τ a mod (∂fτ /∂x). The multiplication • on the tangent spaces is Frobenius with respect to the following residue metric: . . . 1 3 ψa (x)ψb (x)ω . (∂τa , ∂τb )τ := ∂fτ ∂fτ ∂fτ 2π i ∂x1 ∂x2 ∂x3

The residue metric is known to be flat and together with the Frobenius multiplication, the unit vectors ∂τ N and the Euler vector field E :=

N

(deg τ a )τ a ∂τ a ,

deg τ a = 1 − (ma − 1)/ h,

a=1

forms a conformal Frobenius structure on T (see [7]). On the other hand, the condition (∗) involves only the symplectic structure on H and the operator of multiplication by z and thus admits the following twisted loop group of symmetries: L(2) GL(H ) = {M ∈ End(H )((1/z)) | M(−z)∗ M(z) = 1}. According to a result from [14], when the Frobenius structure associated with the cone L is semisimple, one can identify L with the Cartesian product LA1 × · · · × LA1 of N = dim H copies of the cone LA1 defined by the genus 0 descendent potential (0) FA1 = lim→0 ln DA1 . The identification is provided by a certain transformation Mτ from (a completed version of) L(2) GL(H ) whose construction depends on the choice of a semisimple point τ . A number of results in Gromov–Witten theory suggests that the higher genus theory inherits the symmetry group L(2) GL(H ) (see [11, 14]). This motivates the following construction of the total descendent potential of a semisimple Frobenius manifold. Adopt the following rules of quantization ˆ of quadratic Hamiltonians. Let {. . . , pa , . . . , qb , . . . } be a Darboux coordinate system on the symplectic space (H, ) compatible with the polarization H = H+ ⊕ H− . Then


(qa qb )ˆ = qa qb /,

(qa pb )ˆ = qa ∂/∂qb ,

179

(pa pb )ˆ = ∂ 2 /∂qa ∂qb .

This gives a projective representation of the Lie algebra L(2) gl(H ) in the Fock space. The central extension is due to ˆ = {F, G}ˆ + C(F, G), [Fˆ , G] where C is the cocycle satisfying + C(pα pβ , qα qβ ) =

1 if α = β, 2 if α = β

and equal to 0 for any other pair of quadratic Darboux monomials. Introduce the total descendent potential as an asymptotical function: D := C(τ )Mˆ τ [DA1 ⊗ · · · ⊗ DA1 ], where Mˆ := exp(ln M)ˆ, and C(τ ) is a normalizing constant possibly needed to keep the right-hand side independent of the choice of a semisimple point τ . This definition has been tested in [11, 12] and is known to agree with the TRR, SE, DE, and Virasoro constraints. Here is a more explicit description of Mτ and C(τ ) in the form applicable to Frobenius manifolds of simple singularities. Consider the complex oscillating integral efτ (x)/z ω. JB (τ ) = (−2π z)−3/2 B

Here B is a noncompact cycle from the relative homology group lim Hm (Cm , {x : Re(fτ /z) ≤ −c}) ! ZN .

c→∞

We will use the notation ∂1 , . . . , ∂N for partial derivative with respect to a flat (and weighted-homogeneous) coordinate system (t 1 , . . . , t N ) of the residue metric. We treat the derivatives z∂a JB as components of a covector field z ∂a JB dt a ∈ T ∗ T which can be identified with a vector field via the residue metric and—via its LeviCivita connection—with an H -valued function JB (z, τ ). According to K. Saito’s theory, these functions satisfy in flat coordinates the differential equations z∂a J = (∂a •)J

(7)

together with the homogeneity condition (z∂z − µ + z−1 E•)J = 0,

(8)

where µ = −µ∗ is the diagonal operator with the eigenvalues 1/2 − ma / h. The latter equation yields an isomonodromic family of connection operators ∇τ = ∂z − µ/z + (E•)/z2 regular at z = ∞ and turning into ∂z − µ/z at τ = 0.

180


According to [8], there exists a (unique in the ADE case) gauge transformation of the form Sτ (z) = 1 + S1 (τ )z−1 + S2 (τ )z−2 + · · · (i.e., near z = ∞) conjugating ∇τ to ∇0 and such that Sτ∗ (−z)Sτ (z) = 1. It satisfies the homogeneity condition (z∂z + LE )Sτ = [µ, Sτ ]. On the other hand, let τ be semisimple. Then the functions fτ have N nondegenerate critical points x (a) (τ ) with the critical values ua (τ ) and the Hessians a (τ ). The local coordinate system {ua } (called canonical) diagonalizes the product • and the residue metric ∂/∂ua • ∂/∂ub = δab ∂/∂ub ,

(∂/∂ua , ∂/∂ub )τ = δab

Define an orthonormal coordinate system #(τ ) : CN → Tτ T = H,

#(q 1 , . . . , q N ) =

qa

&

−1 b a ∂/∂u .

a ∂/∂u

a

,

and put Uτ = diag[u1 (τ ), . . . , uN (τ )]. Stationary phase asymptotics of the oscillating integrals JBa , a = 1, . . . , N, near the corresponding critical points x (a) yield a fundamental solutions to the system (7), (8) in the form #(τ )Rτ (z)eUτ /z ,

Rτ = 1 + R1 (τ )z + R2 (τ )z2 + · · · +,

Rτt (−z)Rτ (z) = 1.

The matrix series Rτ satisfies the homogeneity condition (z∂z + LE )Rτ = 0 and, according to [11], an asymptotical solution with this property is unique up to reordering or reversing the basis vectors in CN . Define 1 τ aa c(τ ) := R1 (τ )dua 2 a aa a as the local potential of the 1-form R1 du /2 (which is known to be closed [7]). In the above notations, the total descendent potential of the ADE-singularity assumes the form Uˆτ ⊗N D = ec(τ ) Sˆτ−1 #(τ )Rˆ τ e z DA . (9) 1 The right-hand side is known to be independent of τ (see [11]) and defines D (up to a constant factor) as an asymptotical function of q = q0 + q1 z + q2 z2 + · · · in the formal neighborhood of q = τ − z with semisimple τ . Our main result is the following theorem. Theorem 1. The total descendent potential (9) of a simple singularity satisfies the corresponding Hirota quadratic equation (1)–(5). In Section 4, we discuss Hirota quadratic equations of the KdV-hierarchy. The plan for the proof of Theorem 1 is to reduce the Hirota quadratic equations for D to those for DA1 by conjugating the vertex operators in (1), (2) past the quantized symplectic transformations from (9). In Section 5, we describe the results of such conjugations by quoting corresponding theorems from [12]. The residue in (1) is computed in Section 6 and is compared with (2) in Section 7. The case-by-case tables for the coefficients aα are presented in Section 8. A key to all our computations is the phase form and its properties discussed in next section.


181

3 Phase forms and root systems Consider a flat family of cycles φ ∈ H2 (fτ−1 (λ)) in the nonsingular Milnor fibers (0) and define the period vector Iφ (λ, τ ) ∈ H by (0)

(Iφ (λ, τ ), ∂a ) := ∂a

(−1) 2π

φ⊂fτ−1 (λ)

ω . dfτ

(10)

It is a multiple-valued vector function on the complement to the discriminant which (0) turns into Iφ (λ) from Section 1 at τ = 0. ˜ α,β (defined in [12, Section 7]) is given by the formula The phase form W ˜ α,β (λ, τ ) := W

N

(0)

(Iα(0) (λ, τ ) • Iβ (λ, τ ), ∂τ a )dτ a .

i=1

This is a multiple-valued 1-form on the complement to the discriminant and depends bilinearly on the cycles α, β (to be chosen in (f0−1 (1) and transported to fτ−1 (λ)). According to [12], the phase forms have the following properties: ˜ α,β = 0. 1. d W ˜ α,β = 0, i.e., W ˜ is determined by the restriction 2. L∂λ +∂N W ˜ α,β (0, τ ), Wα,β (τ ) := W

˜ α,β (λ, τ ) = Wα,β (τ − λ1). W

3. LE Wα,β = 0. 4. Near a generic point of the discriminant ⊂ T the form Wα,β becomes single(0) valued on the double cover and has a pole of order ≤ 1 on D (since Iα have a pole of order ≤ 1/2). 2 5. δγ Wα,β = −2π iα, γ β, γ , where γ is the cycle vanishing over a generic point of the discriminant, and δγ is a small loop going twice (in the positive direction defined by complex orientations) around the discriminant near this point. Proposition 1. Wα,β = −

1 dγ , x . α, γ β, γ 2 γ , x γ ∈A

Proof. The phase form Wα,β becomes single-valued on the Chevalley cover representing T as the quotient of CN = H 2 (f0−1 (1), C) by the monodromy group. The properties (1) and (4) show that it has at most a logarithmic pole on the mirrors γ , x = 0. Property 5 controls the residues on the mirrors. The difference of the leftand right-hand sides has to be a holomorphic 1-form, homogeneous of degree 0 by property 3 and therefore vanishes identically.

Corollary 1. iE Wα,β = −α, β.

182


Indeed, the Euler vector fieldbecomes h−1 xa ∂xa on the Chevalley cover, so that the equality follows from γ ∈A α, γ β, γ = 2hα, β. This is one more general property of phase forms established in [12]. Corollary 2. The phase form Wβ of Section 1 coincides with Wβ,β . Remark. The inverse to the Chevalley quotient map is given by the period map τ → [ω/dfτ ] ∈ H 2 (fτ−1 (0), C) ; H 2 (f0−1 (1), C) ! CN . (0)

The periods Iα are defined via the differential of the inverse Chevalley map and therefore represent parallel translations of the cycles α considered as covectors in CN . The value of phase form Wα,β , which is also a covector, is constructed as the Frobenius product α • β of covectors (defined by the isomorphisms Tτ T ! Tτ∗ T based on the residue metric). Thus the formula 1 α, γ β, γ γ α • β := 2 γ , x γ ∈A

defines on (CN )∗ a family of commutative associative multiplications depending on the parameter x.5 It would be interesting to find a representation-theoretic interpretation of this structure defined entirely in terms of the root system A. We prove several further properties of phase forms needed in our computations. Proposition 2. In the case of ADE-singularities, suppose that β has integer intersection indices with all α ∈ A and2 is invariant under the monodromy around a discriminant-avoiding loop γ . Then γ Wβ,β ∈ 2π iZ. Proof. This is [12, Section 7, Proposition 1].

It would be interesting to find out if the property remains valid for nonsimple singularities. We will see in Section 7 that the coefficients aα introduced in Section 1 can be equivalently defined via the following limits bα . Start by choosing (τ1 , . . . , τN ) = −1 = (0, . . . , 0, −1) in the role of the base point in T and identify A with the set of −1 vanishing cycles in H2 (f−1 (0)) = H2 (f0−1 (1)). Let us also fix τ ∈ T such that fτ is a Morse function, and let u be one of the critical values of fτ so that τ − u1 ∈ . We may assume that τ − (u + 1)1 ∈ / and that the straight segment connecting τ − (u + 1)1 with τ − u1 does not intersect . For each α ∈ A, pick a discriminantavoiding path γα connecting −1 with τ − (u + 1)1 and further with τ − u1 along the straight segment and such that α becomes the vanishing cycle when transported along γα from 1 to τ − u1. Assuming that integration of the phase form is performed along this path, we put 3 + −ε τ −(u+ε)1 2dt . (11) Wα,α − bα := lim exp − ε→0 t −1 −1 5 We thank V. A. Ginzburg, who explained to us that this is a special case of a family of

Frobenius structures constructed by A. P. Veselov [21].


183

Proposition 3. The limit exists and does not depend on the choice of the path of integration provided that the path terminates at a generic point of the discriminant and that the cycle α transported along the path vanishes over this point. Proof. We may assume that u = u1 is the first of the canonical coordinates U = (u1 , . . . , uN ), and therefore u1 = 0 is the local equation of the discriminant branch. (0) Since α is vanishing at the end of the path, the period vector Iα has the following N expansion (here 1i stand for the standard basis vectors in C ): #τ−1 Iα(0) (λ, τ ) = & Since #(1i ) =

√

±2 2(λ − u1 )

i ∂/∂u

i,

11 + (λ − u1 )

a i (U )1i + o(λ − u1 ) .

we have (1i • 1j , ∂/∂uk ) = δij δik , and therefore

2du1 (Iα(0) • Iα(0) , ∂/∂uk )duk |λ=0 = + 4a 1 (U )du1 + O(−u1 ). −u1 0 u =0 We see that the integral u11=−1 Wα,α diverges the same way as − −1 2dt/t so that the difference converges. This proves the existence of the limit. Removing this singular term we find that the integral [4a1 (U )du1 +O(−u1 )] vanishes along any path inside the discriminant branch u1 = 0. This shows that the limit bα is locally constant as a function of the path’s endpoint on the discriminant and therefore is globally constant due to the irreducibility of the discriminant. Finally, precomposing a path with a discriminant-avoiding loop γ with trivial monodromy of the cycle α does not change bα thanks to Proposition 2.

Wα,α =

Corollary. aα /aβ = bα /bβ for all α, β ∈ A. Proposition 4. Let δε be a small loop of radius ε around the discriminant near a generic point τ − u1, 2 and let α, β = ±1, where β is the cycle vanishing at this point. Then limε→0 δε Wα,α = −π i. Proof. We have α = ±β/2 + α , where α is invariant under the monodromy around (0) (0) (0) δε . Expanding Iα = Iα ± Iβ/2 near λ = u as in the proof of Proposition 3, we find .

. Wα,α = δε

δε

du + −2u

.

√ √ O( u)du = −π i + O( ε) → −π i.

δε

In fact, this property has been already used in [12].

4 Two forms of the KdV-hierarchy Consider the miniversal deformation of the A1 -singularity in the form fu (x) := (x12 + x22 + x32 )/2 + u. The vanishing cycle α can be identified with the real sphere (x12 + x22 + x32 ) = 2(λ − u). The period is

184


& dx1 ∧ dx2 ∧ dx3 d 4 π(2(λ − u))3/2 = 4π 2(λ − u). = dfu dλ 3 α √ (−1) Since (1, 1) = Res dx1 ∧dx2 ∧dx3 /x1 x2 x3 = 1, we have Iα (λ, u) = 2 2(λ − u), (k) and more generally, I±α (λ, u) = ±2(d/dλ)k (2(λ − u))−1/2 , k ∈ Z. The Coxeter transformation swaps α and −α and so aα = a−α = (h + 1)/12h2 = 1/16. The equation (1), (2) in this example assumes the form ( ) dλ A1 ±α 1 A1 ∓α (λ) ⊗ (λ) ( ⊗ ) = 16 l + ( ⊗ ), (12) Resλ=∞ λ 8 ± where l=

2k + 1 2

k≥0

(qk ⊗ 1 − 1 ⊗ qk )(∂qk ⊗ 1 − 1 ⊗ ∂qk ).

(13)

Here we use the notation A1 φ (λ) to single out the vertex operators φ (λ) of the A1 -singularity. In order to identify the condition (12) for with √ the KdV-hierarchy in [16, 17] corresponding to the root system A1 , we denote 2λ by ζ , rescale the + t )/2, y = (t − t )/2, variables by qk = (2k + 1)!! t2k+1 , and put xm = (tm m m m m where m = 1, 3, 5, . . . . In this notation l = mym ∂ym , and (12), (13) becomes 5 4 dζ 4 ζ m √ym −2 ζ −m √∂ym m e e −1−8 mym ∂ym (x + y)(x − y) = 0. Res ζ This coincides with [16, equation (14.13.1)] characterizing tau-functions of the KdV-hierarchy. Another form of the Hirota quadratic equation for is based on the representation of the KdV-hierarchy as the mod 2 reduction of the KP-hierarchy (see [16, Section 14.11]). It can be rephrased (see [12]) as the condition ( ) dλ A1 ∓α/2 A1 ±α/2 (λ) ⊗ (λ) √ ( ⊗ ) has no pole in λ. (14) ± λ ± Indeed, in the previous notations this can be rewritten as the property e

2

ym ζm √ −

e

ζ −m m

√

∂ym

(x + y)(x − y) contains no ζ −m for odd m > 0.

This coincides with the mod 2 reduction of the KP-hierarchy of the Hirota equation [16, equation (14.11.5)]. According to a result from [16, Section 14.13], this condition is actually equivalent to (12). In Section 6, we will use the fact that (according to Kontsevich’s theorem) the function = DA1 satisfies both forms (12) and (14) of the KdV-hierarchy.

5 Symplectic transformations of vertex operators φ

Generalizing the construction of Section 1, introduce the vertex operator τ (λ) corresponding to the vector f ∈ H [[z, z−1 ]] of the form


fτφ (λ) :=

185

(k)

Iφ (λ, τ )(−z)k .

k∈Z (0)

Here Iφ

(k)

is the period vector introduced in Section 3, and Iφ

(0)

:= d k Iφ /dλk as (k)

before. For k < 0, the integration constants are taken “equal to 0’’ so that Iφ satisfy the homogeneity conditions 1 (k) (k) (λ∂λ + LE )Iφ (λ, τ ) = µ − − k Iφ (λ, τ ). 2 φ

In particular, 0 coincides with the vertex operator φ from Section 1. We state below several results about behavior of the vertex operators under conjugation by some symplectic transformations and refer to [12, Sections 5, 6, and 7] for the proofs. Theorem A (see [12, Proposition 2]). φ Sˆτ 0 (λ)Sˆτ−1

+ 3 1 τ −λ1 = exp Wφ,φ τφ (λ). 2 −λ1 φ

We have to stress here that in order to compare the vertex operators 0 (λ) and φ τ (λ), one needs to transport the cycle φ from f0−1 (λ) to fτ−1 (λ) along a path in T connecting −λ1 = (0, . . . , −λ) with τ − λ1 = (τ1 , . . . , τN − λ) and avoiding the discriminant corresponding to singular levels fτ−1 (0). It is assumed in the formulation of the theorem that the integral of the phase form is taken along this very path. Similar conventions apply to other formulas of this and following sections involving integration of phase forms. Now let the cycle φ ∈ H2 (fτ−1 (λ) be written as the sum φ = φ, ββ/2 + φ , where φ , β = 0. Here β is the cycle vanishing at a nondegenerate critical point of the function fτ with the critical value u and transported to fτ−1 (λ) along a discriminantavoiding path connecting τ − λ1 and τ − u1. Theorem B (see [12, Proposition 4]). 3 + τ −u1 φ,β φ, β β Wβ,φ τφ (λ)τ 2 (λ). τφ (λ) = exp 2 τ −λ1 The integral here is taken along the path terminating on the discriminant where the phase form is singular. However the singularity is proportional to (λ − u)−1/2 and is therefore integrable. Let us recall that the columns of the matrix Rτ in the asymptotical expansion #(τ )Rτ (z) exp(U/z) correspond to nondegenerate critical points of the Morse function fτ with the critical values ui (τ ). Let βi be the cycle vanishing over ui . Theorem C (see [12, Proposition 3]). 2 cβ (#(τ )Rˆ τ )−1 τcβi (λ)(#(τ )Rˆ τ ) = ec Wi /2 [· · · 1 ⊗ (A1 ui (λ))(i) ⊗ 1 · · · ],

186


where

Wi :=

τ −ui 1 τ −λ1

Wβi ,βi −

τN

2dt N − ui − t N

,

cβ

and A1 u (λ) is the vertex operator of the A1 -singularity with the miniversal deformation

x12 2

+

x22 2

+

x32 2

+ u corresponding to the c-multiple of the vanishing cycle. (0)

The behavior of Iβi near λ = ui is described by the asymptotics 2 (0) # −1 (τ )Iβi (λ, τ ) = & (1i + · · · ), 2(λ − ui ) where 1i is the ith basis vector in CN , and the dots mean higher order powers of λ−ui . Respectively, the vertex operator of the A1 -singularity is more explicitly defined by the series f ∈ C[[z, z−1 ]] of the form f=

dk 2c (−z)k , √ k dλ 2(λ − u) k∈Z

where the branch of the square root should be the same as in the above asymptotics. The subscript (i) indicates the position of the vertex operator in the tensor product operator acting on the Fock space of functions of (q(1) , . . . , q(N ) ) = # −1 (τ )q. The integrand in the formula for Wi considered as a 1-form in the space with coordinates (t 1 , . . . , t N ) identical to parameters of the miniversal deformation, while the notation τ = (τ 1 , . . . , τ N ) is reserved for expressing the limits of integration. The phase form W has a nonintegrable singularity at t = τ − ui 1 which happens to cancel out with that of the subtracted term so that the difference is integrable. Finally, the following result is the special case of Theorem A corresponding to the A1 -singularity. Theorem D (see [12, Proposition 3]). 2 λ 2dt A1 cβ c 0 (λ). e−(u/z)Â1 ucβ (λ) e(u/z)ˆ = exp − 2 λ−ui t In fact, this result can be obtained more directly using Taylor’s formula. Indeed, for any analytic function I (0) , we have ( ) e−u/z I (k) (λ)(−z)k eu/z = I (k) (λ + u)(−z)k , k∈Z

k∈Z

provided that |u| does not exceed the convergence radius of I (0) √ at λ. Thus √ the transformation in the theorem effectively consists in the translation λ − u ; λ along an origin-avoiding path. The integral in the exponent should be taken along this path.


187

6 Residue sum In this section, we compute the residue sum ( ) dλ −α α Resλ=∞ bα 0 (λ) ⊗ 0 (λ) D⊗2 λ

(15)

α∈A

assuming that the coefficients bα are defined as in Proposition 3. Introduce the total ancestor potential ⊗N Aτ := Sˆτ D = ec(τ ) #(τ )Rˆ τ e(Uτ /z)ˆ DA . 1

Applying Theorem A of the previous section, we find that (15) can be rewritten as ( ) Resλ=∞ λdλ cα τα (λ) ⊗ τ−α (λ) A⊗2 (16) τ , α∈A

+ cα = lim exp −

where

ε→0

τ −(u+ε)1 τ −λ1

Wα,α −

−ε −1

2dt t

3 ,

assuming that α ∈ H2 (fτ−1 (λ)) vanishes at λ = u when transported along the path of integration of the phase form. Note that the factor λ−1 dλ in (15) is replaced by λdλ in (16) due to Corollary 1 from Section 3, which shows that + 3 −λ −λ1 dt exp − Wα,α = exp α, α = λ2 . −1 −1 t (g) The ancestor potential Aτ = exp (g−1) Fτ is a tame asymptotical function (g) in the following sense: Fτ considered as a formal function of tka = qka + δk1 δaN satisfies (g)

∂ r Fτ |t=0 = 0 whenever k1 + · · · + kr > 3g − 3 + r. · · · ∂tkarr

∂tka11

⊗N This follows from the analogous property of DA , from the invariance of DA1 under 1 the string flow exp(u/z)ˆ and from the “upper-triangular’’ property of Rˆ τ . We refer to Proposition 5 in [12] for the proof. It is also shown in [12, Section 8] that for tame φ −φ asymptotical functions the vertex operator expressions τ (λ) ⊗ τ (λ)⊗2 can be considered not only as series expansions in fractional powers of λ near λ = ∞, but also as multiple-valued analytical functions defined over the entire range of λ and ramified only on the discriminant. Moreover, the sum in (16) is manifestly invariant under the entire monodromy group (= the ADE-reflection group). Therefore the sum is actually a single-valued differential 1-form on the complement to D. Thus the

188


residue (16) at λ = ∞ coincides with the sum of residues at the critical values λ = ui of the function fτ . Our next goal is to take u = ui and compute the residue. In a neighborhood of λ = u, the monodromy group reduces to Z2 generated by the reflection σ in the hyperplane orthogonal to two vanishing cycles which we denote ±β. First, consider the summand in (16) corresponding to a σ -invariant cycle α ∈ A. (k) The period vectors Iα (λ, τ ) are therefore single-valued analytic functions near λ = τ −λ1 u. In particular, ln cα , which differs from a constant by τ −(u+1)1 Wα,α , is analytic, too. We conclude that λcα τα (λ) ⊗ τ−α (λ)A⊗2 has no pole at λ = u. Next, consider a pair of cycles α± ∈ A transposed by σ and having intersection indices ±1 with β. We have α± = α ± β/2 where σ α = α . We use Theorem B ±β/2 α ±β/2 and then commute τ across # Rˆ exp(U/z)ˆ using to replace τ ± with τα τ Theorems C and D. The terms from (16) corresponding to α = α± turn into

7 6 λdλ τα (λ) ⊗ τ−α (λ) #(τ )Rˆ τ e(Uτ /z)ˆ ⊗ #(τ )Rˆ τ e(Uτ /z)ˆ ⎡ ⎤ ' *(i)

±β/2 ∓β/2 × ⎣· · · 1 ⊗ d± A1 (λ) ⊗ A1 (λ) ⊗ 1 · · · ⎦ D⊗N ⊗ D⊗N . 0

±

A1

0

A1

(17) The coefficients d± here are + . d± = lim exp − ε→0

τ −(u+ε)1 τ −λ1

+

τ −(u+ε)1 τ −λ1

Wα± ,α± −

−ε −1

−ε

Wβ/2,β/2 +

2dt ± t

u−λ

τ −u1 τ −λ1

dt − 2t

−λ u−λ

Wα ,β

dt 2t

3 .

(18)

We have to emphasize that all integrals here except the first one are taken along a short path near λ = u making β vanish, while in the first integral this path is precomposed with a loop transforming α± to β. Let us take λ = u + 1 for the base point for such a loop γ± and rearrange the first integral as − γ±

Wα± ,α± −

τ −(u+ε)1 τ −(u+1)1

Wβ,β +

τ −λ1 τ −(u+1)1

Wα± ,α± .

Combining this with Wα± ,α± = Wα ,α ± Wα ,β + Wβ/2,β/2 , we can rewrite the exponent in (18) as − γ±

Wα± ,α± −

τ −(u+ε)1

τ −(u+1)1 τ −λ1 τ −(u+1)1

Wβ,β −

Wα ,α +

−ε

2dt ± t

−1 τ −(u+ε)1 τ −(u+1)1

τ −(u+ε)1 τ −(u+1)1

Wβ/2,β/2 +

Wα ,β

−ε −1

dt 2t

(19) (20)


−

−ε −1

dt − 2t

u−λ −ε

dt − 2t

−λ u−λ

dt . 2t

189

(21)

−λ The integrals in (21) add up to − −1 dt/2t and contribute λ−1/2 to the coefficients d± . The sum in (20) is a function of λ analytic near λ = u (since α is σ -invariant) and is the same for both cycles α± . The values of (19) may depend on the cycle α± but are independent of λ. We claim that in the limit ε → 0 the difference is an odd multiple of π i. Indeed, transporting α− along the composition γ− γ+−1 yields α+ . On the other hand, 2Wα ,β = Wα2+ ,α+ − Wα− ,α− . Thus the difference of the two values of (19) can be interpreted as Wα− ,α− along a loop γε starting and terminating at τ − (u + ε)1 and transporting α− to α+ . Let us compose it with a small loop δε of radius ε around λ = u. Since α+ transports along this loop back to α− , the composite integral γε δε Wα− ,α− ∈ 2π iZ due to Proposition 2 and does not depend on ε. Our claim therefore follows from Proposition 4. We conclude that d± = ±d0 (λ)λ−1/2 where d0 is a nonvanishing analytic function near λ = u. Now we use the fact that DA1 is a tau-function of the KdV-hierarchy (14) to conclude that the factor in (17) of the form ±

7 dλ 6 ±β/2 ∓β/2 ± √ A1 0 (λ) ⊗ A1 0 (λ) (DA1 ⊗ DA1 ) λ

is everywhere analytic in λ. The same remains true after application of the operator ˆ (U/z)ˆ )⊗2 . The vertex operator τα ⊗ τ−α is analytic near λ = u since α is (# Re σ -invariant. Thus (17) has no pole at λ = u and contributes 0 to the residue sum. Finally, consider the summands in (15) with α = ±β. Applying Theorems C and D, we transform the corresponding summands from (16) to the form ⎡ ⎤ *(i) ' ±β ∓β ⊗2 ⊗2 ⊗2 (#(τ )Rˆ τ e(U/z)ˆ )⊗2 ⎣· · · DA ⊗ eλdλ(A1 0 ⊗ A1 0 )DA ⊗ DA · · ·⎦, 1 1 1 ±

where e = exp −

−ε

−1

2dt − t

u−λ −ε

2dt − t

−λ u−λ

2dt t

= exp −

−λ

−1

2dt t

= λ−2 .

The contribution of these terms to the residue sum (16) at λ = ui can be calculated using the form (12) of the KdV-hierarchy for DA1 and is equal to ˆ (U/z)ˆ )⊗2 l (i) (D⊗N )⊗2 , 16(# Re A1

where l (i) = (· · · 1 ⊗ l ⊗ 1 · · · ).

In order to justify this conclusion, recall from the end of Section 5 that conjugation by exp(ui /z) act as translation λ − ui → λ. Also, since DA1 is tame, the vertex operator expression in (12) yields a meromorphic 1-form in λ with a singularity only at λ = 0. Thus the residue in (12) at λ = ∞ is the same as at λ = 0. Let us summarize our computation.

190


Proposition 5. The residue sum (15) is equal to ' * N N ⊗N ⊗2 c ˆ −1 (U/z)ˆ ⊗2 (i) ˆ (DA 16(e S # Re + ) l ) . 1 8

(22)

i=1

7 The Virasoro operator Functions of the form ⊗ belong to a Fock space which is the quantization of the symplectic space H ⊕ H, the direct sum of two copies of (H, ). Respectively, the operator

ma ∂ ∂ a a + k (qk ⊗ 1 − 1 ⊗ qk ) (23) ⊗1−1⊗ a h ∂qka ∂qk a k≥0

in (2) is the quantization of a certain quadratic Hamiltonian (Df , f )/2 on H ⊕ H. Let us describe the infinitesimal symplectic transformation D explicitly. Introduce the Virasoro operator l0 := z∂z + 1/2 − µ.6 Since µ∗ = −µ, the operator l0 : H → H is antisymmetric with respect to , and the corresponding quadratic Hamiltonian reads as . 1 1 k + − µ fk , (−1)k f−1−k (l0 f (−z), f (z))dz = 4π i 2 k≥0

=−

N ma k≥0 a=1

h

+ k qka pka .

Comparing this with (23), we conclude that 5 4 −l0 l0 ∈ End(H ⊕ H). D= l0 −l0

(24)

The expression (2) on the right-hand side of the Hirota equation is proportional to ˆ Mˆ ⊗2 )(D×N )⊗2 , ˆ ⊗2 = Mˆ ⊗2 (Mˆ ⊗2 )−1 D( DD A1 where Mˆ = ec(τ ) Sˆτ−1 #(τ )Rˆ τ e(Uτ /z)ˆ . Note that Mˆ ⊗2 is the quantization of a blockdiagonal operator 5 4 4 5 −M −1 l0 M M −1 l0 M M 0 −1 . B := and B DB = 0 M M −1 l0 M −M −1 l0 M 6 The name comes from the property of the operators l := l zl z · · · zl (z repeated m times, m 0 0 0

m = −1, 0, 1, 2, . . . ) to form a Lie algebra isomorphic to the algebra of formal vector fields x m+1 ∂/∂x on the line and participating in the formulation of the Virasoro constraints (see [11, 14]).


Proposition 6. M −1 l0 M =

N

i=1 (

A1 l

0)

191

(i) .

Proof. We have E• 1 1 S z∂z + − µ S −1 = z∂z + − µ + , 2 2 z since (z∂z +LE )S = µS−Sµ and ∂a S = z−1 ∂a •S. Next, in the canonical coordinates, E = ui ∂/∂ui , and therefore E• U 1 1 −1 # z∂z + − µ + # = z∂z + − V + , 2 z 2 z where V := # −1 µ# = # −1 LE #. Furthermore, the differential equations ∂a (#ReU/z ) = z−1 (∂a •)(#ReU/z ) translate into (d + # −1 d#)R = z−1 (dU R − RdU ). This implies (LE + V )R = z−1 (U R − RU ), which together with the homogeneity condition (z∂z + LE )R = 0 shows that U 1 1 U R −1 z∂z + − V + R = z∂z + + . 2 z 2 z Finally, e

−U/z

1 U z∂z + + 2 z

1 eU/z = z∂z + . 2

Proposition 7. Mˆ −1 lˆ0 Mˆ = (M −1 l0 M)ˆ+ tr µµ∗ /4. Proof. The quadratic Hamiltonians for z∂z + 1/2, µ, V , ln S, (E•)/z, U/z contain no p 2 -terms, and the quadratic Hamiltonians for z∂z + 1/2, µ, V , ln R contain no q 2 -terms. Therefore, in the quantized version of the previous computation, the only point where the cocycle C makes a nontrivial contribution is U U Rˆ −1 ˆRˆ = R −1 R ˆ + C. z z Let A = ln R, B = U/z. Then the quadratic Hamiltonian of BA − AB contains no q 2 -terms (since R|z=0 = 1). We therefore have d −t Aˆ ˆ t Aˆ ˆ ˆ t Aˆ = e−t Aˆ (BA − AB)êt Aˆ + C(B, A) e Be = e−t A (Bˆ Aˆ − Aˆ B)e dt 6 7 d 6 −tA tA 7 = e−tA (BA − AB)etA ˆ + C(B, A) = e Be ˆ + C(B, A). dt Integrating in t from 0 to 1 wefind C = C(B, A). Since A = R1 z + o(z), we compute explicitly C = tr(BA)/2 = i R1ii ui /2.

192


This expression, which seems to be a function of τ , has to be a constant, and the value of this constant is well known to be tr µµ∗ /4 (see, for instance, the last chapter in [15]). For the sake of completeness, we include the computation. Namely, comparing the z0 - and z1 -terms in the equation (LE + V )R = z−1 (U R − RU ) we ij find V ij = (ui − uj )R1 and, respectively, R1ii = −LE R1ii =

V ij V j i ij j i (ui − uj )R1 R1 = . uj − u i j

j

Thus we have uj V ij V j i 1 i ii ui V ij V j i 1 ij j i 1 = =− u R1 = V V = tr µµ∗ , j i i j 2 2(u − u ) 2(u − u ) 4 4 i

ij

ij

ij

since V = # −1 µ# and V t = # −1 µ∗ #.

Remark. Slightly generalizing Propositions 6 and 7, one obtains the following trans (i) formation formula (see Theorem 8.1 in [11]) Mˆ −1 lˆm Mˆ = i A1 lˆm for the Virasoro ˆ ⊗N operators with m = 0. Since (lˆm − δm,0 /16)DA1 = 0, this implies that D = MD A1

satisfies the Virasoro constraints [lˆm − δm,0 tr(µµ∗ /4 + 1/16)]D = 0. In fact, this is [11, Corollary 8.2] specialized to Frobenius structures of weighted-homogeneous singularities. Note that the conjugation l0 → M −1 l0 M of the off -diagonal blocks in the matrix D yields after quantization Mˆ −1 lˆ0 Mˆ = (M −1 l0 M)ˆ (since the cocycle C vanishes on pairs of quadratic Hamiltonians corresponding to block-diagonal and block-off diagonal operators.) Thus Bˆ −1 Dˆ Bˆ = i l (i) − tr µµ∗ /2. Taking into account that 1 1 1 N (h + 1) ma (h − ma ) = + µ − µ = a a 12h 2 a 2 2 2h2 a 1 1 = tr + µµ∗ , 2 4 we conclude that the right-hand side of the Hirota equation (1), (2) can be written as ' * N ⊗N ⊗2 ⊗2 (i) (DA + l ) . Mˆ 1 8 i

Comparing this with Proposition 5, we arrive at the following result. Proposition 8. The function D satisfies the Hirota quadratic equation (1), (2) with aα = bα /16. Since D = 0, the Hirota equation is thus rendered consistent, and the following corollary completes the proof of Theorem 1.


193

Corollary. The average value 4(h + 1) 1 bα = . Nh 3h2 α∈A

Note that in the proof of Theorem 1, we use neither the Virasoro constraints for ⊗N DA1 nor the fact that the N factors in DA are the same. The only relevant conditions 1 for DA1 were both forms of the KdV-hierarchy and the tame property of exp(u/z)ˆDA1 . Thus we have actually proved the following generalization of Theorem 1. Theorem 2. Suppose that tame asymptotical functions 1 , . . . , N are tau-functions of the KdV-hierarchy and remain tame under the string flow i → exp(u/z)î for all u. Then := ec(τ ) Sˆτ−1 #(τ )Rˆ τ e(Uτ /z)ˆ (1 ⊗ · · · ⊗ N ) satisfies the corresponding Hirota quadratic equation (1)–(5). Remark. Although the condition for i to remain tame under the string flow is quite restrictive, DA1 is not the only tau-function satisfying it. A large class of examples consists of the shifts DA1 (q + a) where a(z) = a0 + a1 z + a2 z2 + · · · is a series with coefficients ak which are arbitrary series in such that a0 and a1 are smaller than 1 in the -adic norm and ak → 0 in this norm as k → ∞.

8 Kac–Wakimoto hierarchies Let us compare theADE-hierarchies (1)–(5) with the principal hierarchies of the types (1) (1) (1) AN , DN , EN described in [17, Theorem 1.1]. The corresponding Hirota equation [17, equation (1.14)] has the form dζ m∈E 2βi,m −1/2 ym ζ m −m∈E βi,−m 1/2 ∂ym ζ −m /m + + gi e e (x + y)(x − y) ζ i=1 ⎞ ⎛ (25) mym + ρ, ρ⎠ (x + y)(x − y). = ⎝2h N

Res

m∈E+

Here ρ is the sum of the fundamental weights of the root system A, and the value ρ, ρ = Nh(h+1)/12 can be found, for instance, from the tables in [5]. The index set E+ = {ma +kh|a = 1, . . . , N, k = 0, 1, 2, . . . }, and m denote the remainder modulo h. The vertex operators in the sum correspond to a set of roots αi , i = 1, . . . , N, chosen one from each orbit of some Coxeter element M on the root system A. The coefficients βi,m are coordinates of αi with respect to a basis√of eigenvectors Hm of the Coxeter transformation M with the eigenvalues exp(2π −1m/ h) satisfying

194


the additional normalization condition Hm , H−m = 1.7 The coefficients gi are defined via representation theory of affine Lie algebras. The numerical values of gi are computed in [17] in the cases AN , D4 , and E6 . In order to identify the vertex operators in (25) with those in (1), (2) let us start (−1) by taking ζ = (hλ)1/ h . Then the components of the period vector Iαi with respect to a suitable basis [ψa ] ∈ H will have the form ma / h (λ), [ψa ]) = βi,ma m−1 . (Iα(−1) a (hλ) i

(26)

Indeed, the weighted-homogeneous forms ψa ω/df represent a basis of eigenvectors for the classical monodromy operator in H 2 (f −1 (1), C). Then it is straightforward to check that the relation qka =

k 1

(ma + rh)tma +kh

(27)

r=0

(together with the standard change x + y = t , x − y = t as in Section 4) identifies the vertex operators in (25) with αi ⊗ −αi . Note that replacing αi with any of the h roots from the same M-orbit does not change the corresponding residue in (25) since the new vertex operator would differ from the old one only by the choice of the branch of ζ = (hλ)1/ h . Thus we arrive at the following conclusion. Proposition 9. The choice of the basis {[ψa ] ∈ H } such that (26) holds true and the change of variables (27) identify the Hirota equation (1)–(5) with the corresponding hierarchy of the form (25) provided that gi = h3 aαi = h3 bαi /16. Let us now compute the coefficients bα . First, rewrite the definition (11) as bα = lim e

−

τ −(u+ε)1 −ε1

ε→0

Wα,α

= lim

ε→0

1 y(ε), γ γ ∈A

α,γ 2 2

ε 1/ h κ, γ

α,γ 2 2

=

v, α4 κ, α4

1 γ ,α=1

x, γ , κ, γ

where ε1/ h κ, y(ε) and x are inverse images under the Chevalley map of −ε1, τ − (u + ε)1 and τ − u1, respectively, x is a generic point on the mirror α, x = 0, and v is determined from the expansion y(ε) = x + ε1/2 v + o(ε1/2 ). We will use this formula in the case of A and D series. Case AN . The root system consists of the vectors γij := ei − ej in the space CN +1 with the standard orthonormal basis e0 , . . . , eN and coordinates z0 , . . . , zN . Take zN +1 1 1 + t1 zN −1 + · · · + tN = (z − zi ). N +1 N +1 N

F (z, τ ) =

i=0 7 As usual, there is a caveat in the case D with odd l when the eigenvalue −1 of the monl

odromy operator has multiplicity 2. The involution of the Dynkin diagram induces an automorphism of the root system which allows one in this case to single out one invariant and (i) (a) one antiinvariant eigenvector, Hl−1 and Hl−1 , orthogonal to each other and normalized by Hl−1 , Hl−1 = 1 each.


195

Let α = ea − eb and let t = τ − u1 be a generic point on the discriminant. Then the components yi (ε) = xi +ε 1/2 vi +εwi +o(ε) (where xa = xb ) satisfy F (yi , t −ε1) = 0, and therefore ε = F (xi , t) + F (xi , t)ε 1/2 yi + F (xi , t)εwi + F (xi , t)ε

vi2 + o(ε). 2

We have&F (xi , t) = 0 for all i and F (xi , t) = 0 for i = a,& b. This implies that vi = ± 2/F (xa , t) for i = a, b and hence α, v = ±2 2/F (xa , t). Thus α, v4 = 64/F (xa , t)2 . On the other hand, 2 1 1 N −1 2 N −1 (N + 1)F (xa , t) x, γ = (−1) (xi − xa ) = (−1) . 2 i=a,b

γ ,α=1

The eigenvector κ = (N + 1)1/(N +1) (1, η, η2 , . . . , ηN −1 ) of the Coxeter transformation (z0 , . . . , zN ) → (z1 , . . . , zN , z0 ) with the eigenvalue η = exp 2π i/(N + 1) is a preimage of t = −1 under the Chevalley map. We find8 1 1 1 κ, α4 κ, γ = (N + 1)2 (ηa − ηb )2 (ηa − ηj ) (ηi − ηb ) j =a

α,γ =1

i=b

= (−1) (N + 1) (η − η ) η 4

N

b 2 N (a+b)

a

= (−1)N −1 (N + 1)4 (2 − ηa−b − ηb−a ). Collecting the results, we find bα =

1 16 . a−b 2 − ηb−a ) (N + 1) (2 − η

This agrees with [17, Theorem 1.2], where gi = (N + 1)/(2 − ηi − η−i ) corresponds to αi = e0 − ei . In particular,

N + 1 −2 sin gk = 4 N

k=1

πk N +1

=

N (N + 1)(N + 2) . 12

The middle expression is a special case of Dedekind sums, and the second equality, which follows from our results, is well known in number theory (see, e.g., [4]). Case DN . The root system consists of the vectors ±ei ± ej , i = j , where e1 , . . . , eN is the standard orthonormal basis and (z1 , . . . , zN ) are the corresponding coordinates in CN . The parameters (t1 , . . . , tN ) in the following family of polynomials F (z, t) = z2N + t2 z2N−2 + t3 z2N −4 + · · · + tN z2 + t12 =

N 1 (z2 − zi2 )

i=1 8 We use here the facts that the product 8 2π ik/n ) over all nth roots of unity except (ζ − e k=a ζ = e2π ia/n is equal to the derivative of zn − 1 at z = ζ , i.e., to n/ζ .

196


are identified with coordinates on the Chevalley quotient CN /W . Note that the invariant tN of degree h = 2N − 2 is the coefficient at z2 . Let us assume that x is a generic point on the mirror za ± zb orthogonal to the root α = ea ∓ eb , and that t is the corresponding point on the discriminant, so that xa = ±xb and F (±xa , t) = F (±xa , t) = 0. Taking yi (ε) = xi + ε 1/2 vi + εwi + o(ε) and expanding F (y(ε), t1 , . . . , tN − 1, tN − ε) = 0 in ε, we find εxi2 = F (xi , t) + F (xi , t)(ε1/2 vi + εwi ) + F (xi , t)ε

vi2 + o(ε). 2

& & Thus va = 2xa2 /F (xa , t), vb = ∓ 2xa2 /F (xa , t) and α, v4 = 64xa4 /F (xa , t)2 . Furthermore, ⎡ ⎤ 1 1 F (z, t)|z=xa = ⎣2 (z2 − xi2 ) + 4z2 (z2 − xi2 )⎦ a i=a

=

8xa2

1

(xa2

a=b i=a,b

z=xa

− xi2 ).

i=a

Using this we find 1

x, α =

1 j =a,b

α,γ =1

(xa2 − xj2 )

1

(∓1)(xi2 − xb2 ) = (±1)N −2

i=a,b

F (xa , t)2 . 64xa4

Next, the eigenvector κ = (1, η, . . . , ηN −2 , 0) of the Coxeter transformation (z1 , . . . , zN ) → (z2 , . . . , zN −1 , −z1 , zN ) with the eigenvalue η = exp πi/(N − 1) is mapped to (t1 , . . . , tN ) = (0, . . . , 0, 1) under the Chevalley map. Assuming first that α = ea ∓ eb with a, b < N, we find 1 1 κ, γ = (ηa ∓ ηb )4 (ηa )2 (∓ηb )2 (η2a − η2i )(±1)(η2b − η2i ) κ, α4 i=a,b,N

α,γ =1

∓ η b )2 (ηa ± ηb )2 (2 ∓ ηa−b ∓ ηb−a ) . = (±1)N−2 (N − 1)2 (2 ± ηa−b ± ηb−a ) = −(±1)N −2 (N − 1)2

(ηa

Combining with the previous formulas, we compute bα =

(2 ± ηa−b ± ηb−a ) 1 2 (N − 1) (2 ∓ ηa−b ∓ ηb−a )

for α = ea ∓ eb .

Now let α = ea ∓ eN . Then 1 1 κ, γ = η4a (η2a − η2i )(−η2i ) = (−1)N −2 (N − 1) κ, α4 α,γ =1

i=a,N


197

and therefore bα = 1/(N − 1). Taking the representatives α1 = eN −1 − e1 ,

. . . , αN −2 = eN −1 − eN −2 ,

αN −1 = eN −1 − eN ,

αN = eN −1 + eN

in the orbits of the Coxeter transformation on A, we find gi =

(N − 1) (2 − ηi − η−i ) 2 (2 + ηi + η−i )

gi =

(N − 1)2 2

for i = 1, . . . , N − 2

and for i = N − 1, N.

The identity gk = (N − 1)N (2N − 1)/6, which follows from our general theory, agrees with the value of the Dedekind sum9 N −2 k=1

tan

2

πk 2N − 2

=

(N − 2)(2N − 3) . 3

In the case N = 4, the values gi = 1/2, 9/2, 9/2, 9/2 agree with the values of gi found in [17, Proposition 1.3(a)]. Cases EN . We find gi using the packages LiE and MAPLE to compute the ratios via (5) and then apply the normalizing relation (3). In each case EN , let α1 , . . . , αN be the simple roots and M be the Coxeter transformation described by the following diagrams: α 1 α3 α 4 α 5 α 6 • − • − • − • −• | • M = σ1 σ4 σ6 σ2 σ3 σ5 , α2 α1 α 3 α 4 α 5 α 6 α 7 • − • − • − • − • −• | • M = σ1 σ4 σ6 σ2 σ3 σ5 σ7 , α2 α1 α 3 α 4 α 5 α 6 α 7 α8 • − • − • − • − • − • −• | • M = σ 1 σ 4 σ6 σ8 σ 2 σ 3 σ 5 σ 7 . α2 9 It is essentially the same one as in the A-case since sin −2 x − 1 = cot 2 x = tan2 (π/2 − x).

198


One can check (e.g., using LiE) that all simple roots α1 , . . . , αN belong to different M-orbits. The following tables represent the values of the corresponding coefficients gi , while the values of bαi can be obtained from them as in Proposition 9. Case E6 . We have bαi = gi /108, where √ √ g1 = g6 = 16+8 3, g3 = g5 = 16−8 3,

√ g2 = 7+4 3,

√ g4 = 7−4 3.

This agrees with the values of gi found in [17, Proposition 1.3(b)]. Case E7 . We have bαi = 2gi /729. Put u = cos(π/9). Then 27 + 36u + 24u2 , 2 147 g4 = + 12u − 96u2 , 2 21 g6 = − − 48u + 72u2 , 2

g1 =

225 + 36u − 144u2 , 2 9 g5 = − 72u + 72u2 , 2 9 g7 = + 36u + 72u2 . 2 g2 =

g3 =

3 , 2

Case E8 . We have bαi = 2gi /3375. Let u = cos(π/15). Then 33 + 80u + 72u2 − 16u3 , 2 123 g3 = − + 568u + 376u2 − 912u3 , 2 745 g5 = + 584u − 376u2 − 624u3 , 2 35 g7 = − + 156u + 136u2 − 256u3 , 2

g1 =

273 + 132u − 136u2 − 128u3 , 2 109 − 368u − 72u2 + 400u3 , g4 = 2 257 − 1220u − 232u2 + 1376u3 , g6 = 2 19 g8 = − + 68u + 232u2 + 160u3 . 2 g2 =

9 Open questions (a) Formula (9) defines the total descendent potential D as an asymptotical function of q = q0 + q1 z + · · · with semisimple q0 . As shown in [12, Theorem 5], the function DAN extends to arbitrary values of q0 without singularities. We expect the same for DDN and DEN but leave this issue open. (b) B. Dubrovin [7] associates to a Frobenius manifold a dispersionless integrable hierarchy. In particular, the hierarchy (1), (2) for asymptotical functions = exp(F (0) / + F (1) + · · · ) admits the dispersionless limit as → 0 which is an infinite system of equations for F (0) . It is not hard to show that F satisfies the dispersionless hierarchy if and only if the Gaussian distributions := exp{dx2 F(q)/2} (where dx2 F is the quadratic differential of F at x) satisfy the original hierarchy (1), (2) for all x. An elegant explicit characterization in terms of the semiinfinite Grassmannian of those Gaussian distributions which satisfy the hierarchy of the type AN is given in the appendix in [12]. It would be interesting to generalize the characterization to Cases DN , EN .


199

(c) Theorem 1 implies that the genus 0 descendent potential F (0) = lim→0 ln D satisfies the corresponding dispersionless hierarchy. The quadratic forms dx2 F (0) (q) depend only on N parameters τ = τ (x) (due to the property (∗) of the cone L = graph dF (0) ) and have the following explicit description (see the appendix in [12]): τ ([St (z)q(z)]0 • [St (z)q(z)]0 , ∂t a )dt a , 0

a

where [S(z)q(z)]0 = S0 q0 + S1 q1 + · · · denotes the z0 -mode. The corresponding Gaussian distributions therefore satisfy the hierarchy (1)–(5). Taking τ = u1 so that [Sτ q]0 = qk uk /k! we conclude that in particular the hierarchy has the 1-parametric family of Gaussian solutions ⎧ ⎛ ⎞ ⎫ ⎨ 1 u vk vl ⎬ ⎝ = exp qk , ql ⎠ dv . ⎩ 2 0 ⎭ k! l! k≥0

l≥0

This imposes nontrivial constraints on the coefficients aα in the Hirota equation (1). It would be interesting to find out if these constraints are sufficient in order to determine the coefficients unambiguously. (d) Our computations in Section 8 confirm the Conjecture from Section 1 in Cases AN , D4 , E6 and leave it open in Cases DN with N > 4, E7 , and E8 —mostly because the values of the coefficients gi in the Kac–Wakimoto theory remain unknown. A more conceptual approach to the identification of the Hirota equations should rely on the definition of the coefficients gi given in [17] in terms of representation theory. Namely, the vertex operators Ci± ±αi participate in the so-called principal construction of the basis representation of the affine Lie algebra Aˆ N , Dˆ N , or Eˆ N , and gi = Ci+ Ci− . Here Ci± are certain structure constants whose values remain generally speaking unknown. Our successful description of the products Ci+ Ci− via the phase forms suggests that one should look for the intrinsic role of the phase forms in representation theory and for a description of the individual coefficients Ci± in terms of the phase forms or their generalizations. (e) In representation theory, the hierarchies of ADE type form only a part of a larger list of examples including twisted versions of the affine Lie algebras and nonsimply laced Dynkin diagrams. It would be interesting to find the corresponding constructions in singularity theory and, in particular, to associate the Hirota equations with the boundary singularities BN , CN , F4 . (f) B. Dubrovin and Y. Zhang [9] associate an integrable hierarchy to any semisimple Frobenius manifold. In a sense their construction is parallel to the definition (9) of the total descendent potential D (see [11]) and, in particular, yields objects defined in the complement to the caustic. In this regard the vertex operator description of the hierarchies seems more attractive as it is free of this defect. Of course, theADE-hierarchies (1)–(5) are expected to be equivalent to the hierarchies of Dubrovin–Zhang. It would be interesting to confirm this expectation. (g) Conjecturally, the total descendent potential D extends analytically across the caustic values of q0 in the case of K. Saito’s (semisimple) Frobenius structure

200


corresponding to any isolated singularity. (By the way, this is known to be false for boundary singularities or for finite reflection groups other than AN , DN , EN .) Respectively, one should expect the same for the hierarchies of Dubrovin–Zhang. It would be very interesting to give a vertex operator description of the hierarchies together with Theorem 1 for arbitrary (or at least weighted-homogeneous) isolated singularities of functions. The most obvious difficulty is that the vertex operator sum (1) over the set of all vanishing cycles (or even orbits of the classical monodromy operator on this set) becomes infinite beyond the ADE list. Nevertheless we believe that the obstructions can be removed by an appropriate generalization of the concepts involved. The first examples to study here would be the unimodal singularities P8 , X9 , J10 (see [1]). Their miniversal deformations are closely related to the complex crystallographic reflection groups E˜ 6 , E˜ 7 , E˜ 8 (see [19]). Moreover, the question can be extrapolated to the complex crystallographic groups A˜ N , D˜ N , and the threedimensional Frobenius manifold to be called A˜ 1 represents the first challenge. Acknowledgments The authors thank V. Kac and M. Wakimoto for very helpful consultations on the contents of their paper [17], E. Frenkel and P. Pribik for their interest and stimulating discussions, and B. Sturmfels for his recommendation of the LiE package.

References [1] V. I. Arnold, Normal forms of functions near degenerate critical points, Weyl groups Ak , Dk , Ek and Lagrangian singularities, Functional Anal.] Appl., 6-2 (1972), 3–25. [2] V. I. Arnold, S. M. Gousein-Zade, and A. N. Varchenko, Singularities of Differentiable Maps, Vol. II: Monodromy and Asymptotics of Integrals, Monographs in Mathematics, Vol. 83, Birkhäuser, Basel, 1988. [3] S. Barannikov, Quantum periods I: Semi-infinite variations of Hodge structures, Internat. Math. Res. Notices, 2001-23 (2001), 1243–1264. [4] M. Beck, The reciprocity law for Dedekind sums via the constant Ehrhart coefficient, Amer. Math. Monthly, 106-5 (1999), 459–462. [5] N. Bourbaki, Groupes et algèbres de Lie, Hermann, Paris, 1968, Chapters IV–VI. [6] E. Date, M. Jimbo, M. Kashiwara, and T. Miwa, Operator approach to the Kadomtsev– Petviashvili equation: Transformation groups for soliton equations III, J. Phys. Soc. Japan, 50 (1981), 3806–3812. [7] B. Dubrovin, Geometry of 2D topological filed theories, in Integrable Systems and Quantum Groups, Lecture Notes in Mathematics, Vol. 1620, Springer-Verlag, New York, 1996, 120–348. [8] B. Dubrovin. Painlevé transcendents in two-dimensional topological field theory, in The Painlevé Property, CRM Series in Mathematics and Physics, Springer-Verlag, New York, 1999, 287–412. [9] B. Dubrovin and Y. Zhang, Normal forms of hierarchies of integrable PDEs, Frobenius manifolds and Gromov–Witten invariants, arXiv: math.DG/0108160. [10] I. B. Frenkel, Representations of affine Lie algebras, Hecke modular forms and Korteweg–de Vries type equations, in Lie Algebras and Related Topics (New Brunswick, NJ, 1981), Lecture Notes in Mathematics, Vol. 933, Springer-Verlag, Berlin, New York, 1982, 71–110.


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[11] A. Givental, Gromov–Witten invariants and quantization of quadratic hamiltonians, Moscow Math. J., 1-4 (2001), 551–568. [12] A. Givental, An−1 -singularities and nKdV hierarchies, Moscow Math. J., 3 (2003). [13] A. Givental, Asymptotics of the intersection form of a quasi-homogeneous function singularity, Functional Anal. Appl., 16-4 (1982), 294–297. [14] A. Givental, Symplectic geometry of Frobenius structures, Proceedings of the Workshop on Frobenius Structures (MPIM Bonn, July 2002), to appear; arXiv: math.AG/0305409. [15] C. Hertling, Frobenius Manifolds and Moduli Spaces for Singularities, Cambridge Tracts in Mathematics, Cambridge University Press, Cambridge, UK, 2002. [16] V. Kac, Infinite Dimensional Lie Algebras, 3rd ed., Cambridge University Press, Cambridge, UK, 1990. [17] V. Kac and M. Wakimoto, Exceptional hierarchies of soliton equations, Proc. Sympos. Pure Math., 49 (1989), 138–177. [18] M. Kontsevich, Intersection theory on the moduli space of curves and the matrix Airy function, Comm. Math. Phys., 147 (1992), 1–23. [19] E. Looijenga, On the semiuniversal deformation of a simple-elliptic hypersurface singularity, Topology, 17 (1977), 23–40. [20] K. Saito, On a linear structure of the quotient variety by a finite reflection group, Publ. Res. Inst. Math. Sci., 29-4 (1993), 535–579. [21] A. P. Veselov, On generalizations of Calogero–Moser–Sutherland quantum problem and WDVV equations, J. Math. Phys., 43-11 (2002), 5675–5682. [22] E. Witten, Two-dimensional gravity and intersection theory on moduli space, Surv. Differential Geom., 1 (1991), 243–310.

Momentum maps and measure-valued solutions (peakons, filaments, and sheets) for the EPDiff equation∗ Darryl D. Holm1,2 and Jerrold E. Marsden3 1 Computer and Computational Science Division

Los Alamos National Laboratory MS D413 Los Alamos, NM 87545 USA [email protected] 2 Mathematics Department Imperial College London SW7 2AZ UK [email protected] 3 Control and Dynamical Systems 107-81 California Institute of Technology Pasadena, CA 91125 USA [email protected] To Alan Weinstein on the occasion of his 60th birthday. Abstract. This paper is concerned with the dynamics of measure-valued solutions of the EPDiff equations, standing for the Euler–Poincaré equations associated with the diffeomorphism group (of Rn or of an n-dimensional manifold M). It focuses on Lagrangians that are quadratic in the velocity fields and their first derivatives, that is, on geodesic motion on the diffeomorphism group with respect to a right invariant Sobolev H 1 metric. The corresponding Euler–Poincaré (EP) equations are the EPDiff equations, which coincide with the averaged template matching equations (ATME) from computer vision and agree with the Camassa–Holm (CH) equations for shallow water waves in one dimension. The corresponding equations for the volume-preserving diffeomorphism group are the LAE (Lagrangian averaged Euler) equations for incompressible fluids. ∗ The first author is grateful for support by US DOE under contract W-7405-ENG-36 for Los

Alamos National Laboratory, and Office of Science ASCAR/AMS/MICS. The research of the second author was partially supported by the California Institute of Technology, by the National Science Foundation through NSF grant DMS-0204474, and by Air Force contract F49620-02-1-0176.

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D. D. Holm and J. E. Marsden

It is shown that the EPDiff equations are generated by a smooth vector field on the diffeomorphism group for sufficiently smooth solutions. This is analogous to known results for incompressible fluids—both the Euler equations and the LAE equations—and it shows that for sufficiently smooth solutions, the equations are well posed for a short time. Numerical evidence suggests that as time progresses these smooth solutions break up into singular solutions which, at least in one dimension, exhibit soliton behavior. These nonsmooth, or measure-valued, solutions are higher-dimensional generalizations of the peakon solutions of the CH equation in one dimension. One of the main purposes of the paper is to show that many of the properties of these measure-valued solutions can be understood by the fact that their solution Ansatz is a momentum map. Some additional geometry is also pointed out, for example, that this momentum map is one part of a dual pair.

1 Introduction This paper is concerned with solutions of the EPDiff equations, that is, with the Euler–Poincaré equations associated with the diffeomorphism group in n-dimensions. In particular, we are concerned with singular solutions that generalize the peakon solutions of the Camassa–Holm (CH) equation from one dimension to more spatial dimensions. The CH equation (see Camassa and Holm [1993]) for the dynamics of shallow water in a certain asymptotic regime,1 is ut + 3uux = α 2 (uxxt + 2ux uxx + uuxxx ),

(1.1)

where u(x, t) is the fluid velocity, subscripts denote partial derivatives in position x and time t, α 2 is a positive constant, and the linear dispersion terms normally in CH have been omitted. Equivalently, in Hamiltonian form, this dispersionless CH equation reads as mt = −umx − 2ux m = {m, h(m)}, (1.2) where m = u − α 2 uxx and α 2 is a positive constant. As Camassa and Holm [1993] show, the CH equation is expressed in Hamiltonian form by using the Lie–Poisson bracket {·, ·} defined on the dual Lie algebra of the one-dimensional vector fields and using the Hamiltonian 1 h(m) = umdx. (1.3) 2 The CH equation may be equivalently expressed in Euler–Poincaré form by using the Lagrangian associated with the H 1 metric for the fluid velocity. This Lagrangian is given as a function of the fluid velocity by the quadratic form 1 (1.4) l(u) = (u2 + α 2 u2x )dx. 2 It follows from Euler–Poincaré theory (see Marsden and Ratiu [1999] and Holm, Marsden, and Ratiu [1998a]) that the one-parameter curve of diffeomorphisms η(x0 , t) depending on parameter t and defined implicitly by 1 See Dullin, Gottwald, and Holm [2001, 2003, 2004] for recent discussions of the derivation

and asymptotic validity of the CH equation for shallow water waves, at one order beyond the Korteweg–de Vries equation.

Measure-valued momentum map

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∂ η(x0 , t) = u(η(x0 , t), t) ∂t is a geodesic in the group of diffeomorphisms of R (or, with periodic boundary conditions, of the circle S 1 ) equipped with the right invariant metric equal to the H 1 metric at the identity. A remarkable analytical property of the CH equation, conjectured by keeping track of derivative losses in Holm, Marsden, and Ratiu [1998a] and proved in Shkoller [1998] is that the geodesic equations literally define a smooth vector field in the Sobolev H s topology for s > 3/2. That is, in the material representation, the equations have no derivative loss. This property is analogous to the corresponding results for the Euler equations for ideal incompressible fluid flow (discovered by Ebin and Marsden [1970]) and the Lagrangian averaged Euler equations (again conjectured by Holm, Marsden, and Ratiu [1998a] and proved by Shkoller [1998]). As we will explain in Section 3, a similar statement holds for the n-dimensional EPDiff equation if we use the H 1 metric. This is all the more remarkable because smoothness of the geodesic flow is probably not true for the L2 metric. Smoothness of volume-preserving geodesic flow with respect to the L2 metric does hold for the incompressible flow of an ideal Euler fluid, a result proved in Ebin and Marsden [1970]. Before proceeding with a discussion of the general case of the n-dimensional EPDiff equations, we shall quickly review, mostly to establish notation, a few facts about the Euler–Poincaré and Lie–Poisson equations, whose basic theory is explained, for example, in Marsden and Ratiu [1999]. Review of Euler–Poincaré and Lie–Poisson equations Let G be a Lie group and g its associated Lie algebra (identified with the tangent space to G at the identity element), with Lie bracket denoted [ξ, η] for ξ, η ∈ g. Let : g → R be a given Lagrangian and let L : T G → R be the right invariant Lagrangian on G obtained by translating from the identity element to other points of G via the right action of G on T G. A basic result of Euler–Poincaré theory is that the Euler–Lagrange equations for L on G are equivalent to the (right) Euler–Poincaré equations for on g, namely, to d δ δ = − ad ∗ξ . dt δξ δξ

(1.5)

Here ad ξ : g → g is the adjoint operator, that is, the linear map given by the Lie bracket η → [ξ, η] and ad ∗ξ : g∗ → g∗ is its dual, that is, ad ∗ξ (µ), η = µ, [ξ, η], where , denotes the natural pairing between g∗ and g. Also, δ/δξ denotes the functional derivative of with respect to ξ ∈ g; it is defined to be the element of g∗ such that Dl(ξ ) · η = δl/δξ, η for all η ∈ g, where D denotes the (Frechet) derivative.2 For left invariant systems, we change the sign of the right-hand side in 2 Of course in the finite-dimensional case there is no real difference between Dl and δl/δξ , but in the infinite-dimensional case one normally does not choose g∗ to be the naive, that

is, the literal functional analysis dual, but rather a convenient space for PDE needs.

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(1.5). The Euler–Poincaré equations can be written in the variational form δ dt = 0,

(1.6)

for all variations of the form δξ = η˙ − [ξ, η] for some curve η in g that vanishes at the endpoints. If the reduced Legendre transformation ξ → µ = δ/δξ is invertible, then the Euler–Poincaré equations are equivalent to the (right) Lie–Poisson equations µ˙ = − ad ∗δh/δµ µ,

(1.7)

where the reduced Hamiltonian is given by h(µ) = µ, ξ − (ξ ). These equations are equivalent (via Lie–Poisson reduction and reconstruction) to Hamilton’s equations on T ∗ G relative to the Hamiltonian H : T ∗ G → R, obtained by right translating h from the identity element to other points via the right action of G on T ∗ G. The Lie–Poisson equations may be written in the Poisson bracket form F˙ = {F, h},

(1.8)

where F : g∗ → R is an arbitrary smooth function and the bracket is the (right) Lie–Poisson bracket given by 4 5 δF δG , {F, G}(µ) = µ, . (1.9) δµ δµ In the important case when is quadratic, the Lagrangian L is the quadratic form associated to a right invariant Riemannian metric on G. In this case, the Euler– Lagrange equations for L on G describe geodesic motion relative to this metric and these geodesics are then equivalently described by either the Euler–Poincaré, or the Lie–Poisson equations. Outline of the paper The main contents of this paper are as follows: 1. In Section 2 we review some basic facts about the EPDiff equations, and in particular we recall a singular solution ansatz of Holm and Staley [2003, 2004] (see equation (2.8) below) which introduces a class of singular solutions that generalize the peakon solutions of the CH equation to higher spatial dimensions. 2. In Section 3 we show that the EPDiff equations possess an interesting smoothness property, namely, they define a smooth vector field (that is, they define ODEs with no derivative loss) in the Lagrangian representation. There are a number of interesting consequences of this; in particular, it implies that the EPDiff equations are locally well posed for sufficiently smooth initial data and that the H 1 diameter of


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Diff (M) is strictly positive. Because of the development of singularities in finite time, which the numerics suggests, the smooth solutions may not exist globally in time. This smoothness property is similar to the corresponding smoothness property of the Euler equations for ideal incompressible fluid mechanics shown in Ebin and Marsden [1970]. 3. In Section 4, we show that the singular solution ansatz—again see (2.8) below— defines an equivariant momentum map. We do this in a natural way by identifying the singular solutions with certain curves in the space of embeddings Emb(S, Rn ) of a generally lower-dimensional manifold S into the ambient space Rn (or an n-manifold M) and letting the diffeomorphism group act on this space. The right action of Diff (S) corresponds to the right invariance of the EPDiff equations, while the left action of Diff (Rn ) has a momentum map that gives the desired solution ansatz. This is the main result of the paper. 4. In Section 5 we briefly explore some of the geometry of the singular solution momentum map, in parallel with the corresponding work on singular solutions (vortices, filaments, etc.) for the Euler equations of an ideal fluid that was developed in Marsden and Weinstein [1983]. 5. Finally, in Section 6, we discuss some of the remaining challenges and speculate on some of the many possible future directions for this work. Historical note This paper is dedicated to our friend and collaborator Alan Weinstein and, for us, this work parallels some of our earlier collaborations with him. Alan’s basic works on reduction, Poisson geometry, semidirect product theory, and stability in mechanics— just to name a few areas—have been, and remain, incredibly influential and important to the field of geometric mechanics. See, for instance, Marsden and Weinstein [1974], Weinstein [1983b], Marsden, Ratiu, and Weinstein [1984], Weinstein [1984], and Holm et al. [1985]. Mechanics on Lie groups was pioneered by Arnold [1966], a reference that is a key foundation for the subject and in particular for this paper. However, this theory was in a relatively primitive state, even by 1980, and it has benefited greatly from Alan’s insights. In fact, the clear distinction between the Euler–Poincaré and Lie– Poisson equations, the former equations on g and possessing a variational structure (with constraints on the variations) and the latter on g∗ with its Lie–Poisson structure took until the 1980s to crystallize, and for the place of Lie and Poincaré in the history of the subject to be clarified. This development and clarification was greatly aided by Alan’s work, historical researches, and deep insight. Alan has made key contributions to many fundamental concepts in geometric mechanics, such as Lagrangian submanifolds and related structures (Weinstein [1971, 1977]), symplectic reduction (Marsden and Weinstein [1974]), normal modes and periodic orbits (Weinstein [1973, 1978]), Poisson manifolds (Weinstein [1983b]), geometric phases (Weinstein [1990]), Dirac structures (Courant and Weinstein [1988]) groupoids and Lagrangian reduction (Weinstein [1996]) and the plethora of related “oid’’ structures he has been working on during the last decade (just look over the

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151+ papers on MathSciNet he has written!) that will surely play as an important role in the next generation of people working in the area of geometric mechanics as it is with the current new generation. Of Alan’s papers, the one that is most directly relevant to the topics discussed in this paper is Marsden and Weinstein [1983]. Alan himself is still developing the mathematics associated with this area, as in Weinstein [2002].

2 The EPDiff equation This section reviews the EPDiff equation; that is, the Euler–Poincaré (EP) equation associated with the diffeomorphism group of an n-manifold M (which, for simplicity, will be taken primarily as Rn ). This equation coincides with the dispersionless case of the CH equation for shallow water waves in one and two dimensions, discussed in Camassa and Holm [1993]; Kruse, Scheurle, and Du [2001]. It also coincides with the ATME equation (the averaged template matching equation) in two dimensions. The latter equation arises in computer vision; see, for instance, Mumford [1998], Hirani, Marsden, and Arvo [2001], or Miller, Trouvé, and Younes [2002] for a description and further references. We have chosen to call this by a generic name, the EPDiff equation, because it has these various interpretations in different applications. Of course these different interpretations also provide opportunities: for example, this point of view may enable one to see to what extent the singular solutions found in the EPDiff equations are applicable, either for shallow water wave interactions, or for computer vision applications. A recent combination of these ideas in which image processing is informed by concepts of momentum originating in soliton theory appears in Holm, Trouvé, Ratnanather, and Younes [2004]. Statement of the EPDiff equations Treating analytical issues formally at this point, let X denote the Lie algebra of vector fields on an n-dimensional manifold M (such as Rn ). The space X is the algebra of the diffeomorphism group of M, but the usual Jacobi–Lie bracket is the negative of the (standard) Lie algebra bracket. (See Marsden and Ratiu [1999] for a discussion.) Let : X → R be a given Lagrangian and let M denote the space of oneform densities on M, that is, the momentum densities. The corresponding momentum density of the fluid is defined as m=

δ ∈ M, δu

which is the functional derivative of the Lagrangian with respect to the fluid velocity u ∈ X. If u is the basic dynamical variable, the EPDiff equations are simply the Euler– Poincaré equations associated with this Lagrangian. Equivalently, if m is taken to be the basic dynamical variable, the Legendre transformation allows one to identify the EPDiff equations as the Lie–Poisson equations associated with the resulting


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Hamiltonian. For the case of Rn , we will use vector notation for the momentum density m(x, t) : Rn × R → Rn (a bold m instead of a lightface m). The EPDiff equations are as follows (see Holm, Marsden, and Ratiu [1998a,b]; Holm et al. [2002] for additional background and for techniques for computing the Euler–Poincaré equations for field theories), ∂ T m + 9u ·:; ∇m< + 9∇u:; · m< + m(div u) = 0. (2.1) 9 :; < ∂t convection

stretching

expansion

In coordinates i = 1, 2, . . . , n, using the summation convention, and writing m = mi dx i ⊗ d n x (regarding m as a one-form density) and u = ui ∂/∂x i (regarding u as a vector field), the EPDiff equations read xi ,

∂mi ∂uj ∂uj ∂ mi + uj j + mj i + mi j = 0. ∂t ∂x ∂x ∂x The EPDiff equations can also be written concisely as

(2.2)

∂m + £u m = 0, (2.3) ∂t where £u m denotes the Lie derivative of the momentum one-form density m with respect to the velocity vector field u. As mentioned earlier, if is a quadratic function of u, then the EPDiff equation (2.1) or, equivalently, (2.3), is the Eulerian description of geodesic motion on the diffeomorphism group of the underlying space (in this case Rn ). The corresponding metric is the right invariant metric on the group, whose value on the Lie algebra (the group’s tangent space at the identity—the space of vector fields) is defined by . Since the Lagrangian is positive and quadratic in u, the momentum density is linear in u and so defines a positive symmetric operator Qop by δ = Qop u. δu Likewise, for quadratic Lagrangians the velocity u is determined from the momentum m by u = G ∗ m, where G∗ represents convolution with the Green’s function G for the linear operator Qop . m=

Variational formulation Following the variational formulation of EP theory, the particular EP equation (2.1) may be derived from the following constrained variational principle: δ (u)dt = 0. The variations are constrained to have the form ˙ + w · ∇u − u · ∇w. δu = w This assertion may of course be verified directly. These constraints are analogous to the so-called “Lin constraints’’ used for a similar variational principle for fluid mechanics. (See Marsden and Ratiu [1999] for a discussion and references.)

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Hamiltonian formulation The Legendre transformation yields the Hamiltonian H (m) = m, u − (u), where , is the natural pairing between one-form densities and vector fields given by integration (L2 pairing). This Hamiltonian is the corresponding quadratic form for the momentum, namely, H (m) = (Q−1 (2.4) op (m)). Of course it often happens that Qop is a differential operator and in this case the inverse is usually given in terms of the convolution with the Green’s function G, corresponding to the appropriate solution domain and boundary conditions: u=

δH (m) = G ∗ m. δm

According to the general theory, the EP equation (2.1) may be expressed in Hamiltonian form by using the Lie–Poisson bracket on M as ∂ m = {m, H }LP = − ad ∗δH /δm m. ∂t

(2.5)

One-dimensional CH peakon solutions We return now to the CH equation (1.2), which, as we have noted, is the same as the EPDiff equation (2.1) for the case of one spatial dimension when the momentum velocity relationship is defined by the Helmholtz equation, m = u − α 2 uxx . In one dimension, the CH equation has solutions whose momentum is supported at points on the real line via the following sum over Dirac delta measures: m(x, t) =

N

pi (t)δ(x − qi (t)).

(2.6)

i=1

The velocity corresponding to this measure-valued momentum is obtained by convolution u = G ∗ m with the Green’s function, G(|x − y|) = 12 e−|x−y|/α , for the one-dimensional Helmholtz operator, Qop = (1 − α 2 ∂x2 ), appearing in the CH momentum velocity relationship m = Qop u. Consequently, the CH velocity corresponding to this momentum is given by a superposition of peaked traveling wave pulses, N 1 u(x, t) = pi (t)e−|x−qi (t)|/α . (2.7) 2 i=1


211

Thus the superposition of “peakons’’in velocity arises from the delta function solution ansatz (2.6) for the momentum. Remarkably, the isospectral eigenvalue problem for the CH equation implies that only these singular solutions emerge asymptotically in the solution of the initial value problem in one dimension, as is shown in Camassa and Holm [1993]. Figure 2.1 shows the emergence of peakons from an initially Gaussian velocity distribution and their subsequent elastic collisions in a periodic one-dimensional domain.3 This figure demonstrates that singular solutions dominate the initial value problem. Thus it is imperative to go beyond smooth solutions for the CH equation; as we shall see, there is numerical evidence that the situation is similar for the EPDiff equation.

Fig. 2.1. This figure shows a smooth localized (Gaussian) initial condition for the CH equation breaking up into an ordered train of peakons as time evolves (the time direction being vertical, which then eventually wrap around the periodic domain and interacting with other slower emergent peakons and causing a phase shift (see Alber and Marsden [1992]).

Remarkably, the dynamical equations for pi (t) and qi (t), i = 1, . . . , N, that arise from solution ansatz (2.6)–(2.7) comprise an integrable system for any N . This system is studied in (Alber, Camassa, Fedorov, Holm, and Marsden [2001]) and references therein. See also Vaninsky [2002, 2003] for discussions of how the integrable dynamical system for N peakons is related to the Toda chain with open ends. Generalizing the CH peakon solutions to n dimensions Building on the peakon solutions for the CH equation and the pulsons for its generalization to other traveling-wave shapes (see Fringer and Holm [2001]), the papers of Holm and Staley [2003, 2004] introduced the following measure-valued (that is, density valued) ansatz for the n-dimensional solutions of the EPDiff equation (2.1): m(x, t) =

N

Pa (s, t)δ(x − Qa (s, t))ds.

a=1 3 Figure 2.1 was kindly supplied by Martin Staley.

(2.8)

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These solutions are vector-valued functions supported in Rn on a set of N surfaces (or curves) of codimension (n − k) for s ∈ Rk with k < n. They may, for example, be supported on sets of points (vector peakons, k = 0), one-dimensional filaments (strings, k = 1), or two-dimensional surfaces (sheets, k = 2) in three dimensions. One of the main results of this paper is the theorem stating that the singular solution ansatz (2.8) is an equivariant momentum map. This result helps to organize the theory and to suggest new avenues of exploration, as we shall explain. Substitution of the solution ansatz (2.8) into the EPDiff equations (2.1) implies the following integro-partial-differential equations (IPDEs) for the evolution of such strings and sheets, ∂ a Q (s, t) = ∂t N

b=1

∂ a P (s, t) = − ∂t N

Pb (s , t)G(Qa (s, t) − Qb (s , t))ds ,

(Pa (s, t) · Pb (s , t))

b=1

∂ ∂Qa (s, t)

(2.9)

G(Qa (s, t) − Qb (s , t))ds .

Important for the interpretation of these solutions, the coordinates s ∈ Rk turn out to be Lagrangian coordinates. The velocity field corresponding to the momentum solution ansatz (2.8) is given by u(x, t) = G ∗ m =

N

Pb (s , t)G(x − Qb (s , t))ds ,

u ∈ Rn .

(2.10)

b=1

When evaluated along the curve x = Qa (s, t), the velocity satisfies N u(x, t)x=Qa (s,t) =

Pb (s , t)G(Qa (s, t) − Qb (s , t))ds =

b=1

∂Qa (s, t) . (2.11) ∂t

Thus the lower-dimensional support sets defined on x = Qa (s, t) and parameterized by coordinates s ∈ Rk move with the fluid velocity. Moreover, equations (2.9) for the evolution of these support sets are canonical Hamiltonian equations, δHN ∂ a Q (s, t) = , ∂t δPa

∂ a δHN P (s, t) = − a . ∂t δQ

(2.12)

The Hamiltonian function HN : (Rn × Rn )N → R is 1 HN = 2

N

(Pa (s, t) · Pb (s , t))G(Qa (s, t) − Qb (s , t))dsds .

(2.13)

a,b=1

This is the Hamiltonian for geodesic motion on the cotangent bundle of a set of curves Qa (s, t) with respect to the metric given by G. This dynamic was investigated numerically in Holm and Staley [2003, 2004] to which we refer for more details of the solution properties.


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As we have mentioned, one of our main goals is to show that the solution ansatz (2.8) can be recast in terms of an equivariant momentum map that naturally arises in this problem. This geometric feature underlies the remarkable reduction properties of the EPDiff equation and “explains’’ why the preceding equations must be Hamiltonian—it is because it is a general fact that equivariant momentum maps are Poisson maps. As explained in general terms in Marsden and Weinstein [1983], the way one implements a coadjoint orbit reduction is through a momentum map, and this holds even for the case of singular orbits (again ignoring functional analytic details). Thus, in summary, the Ansatz (2.12) is the EPDiff analog of the corresponding Anzatz for incompressible fluid mechanics (that is, the EPDiffVol equations) that gives point (or blob) vortex dynamics, vortex filaments, or sheets. There are, however, some important differences between vortex dynamics for incompressible flows and the dynamics of the measure-valued EPDiff momentum solutions. For example, the Lagrangian representations of the equations of motion show that EPDiff solutions for momentum have inertia, while the corresponding solutions for point (or blob) vortices of the EPDiffVol dynamics have no inertia. What this means is the following: the equations of motion for the spatial vectors specifying the measure valued vorticity solutions on EPDiffVol are first order in time, while the dynamical equations for the corresponding spatial vectors Qa (s, t) for measurevalued momentum solutions on EPDiff are second order in time. This difference has profound effects on the properties of the solutions, especially on their stability properties. Numerical investigations of Holm and Staley [2003, 2004] show, for example, that the codimension-one singular momentum solutions of EPDiff are stable, while its higher-codimension singular momentum solutions are very unstable to codimensionone perturbations. In contrast, the codimension-two singular vorticity solutions of EPDiffVol (point vortices in the plane, and vortex filaments in space) are known to be stable to such perturbations. Comments on the physical meaning of the equations The EPDiff equations with the Helmholtz relation between velocity and momentum are not quite the CH equations for surface waves in 2D. Those would take precisely the same form, but the shallow water wave relation in the 2D CH approximation would be m = u − α 2 Grad Div u,

that is,

mi = ui − α 2 uj,j i ,

that is,

mi = ui − α 2 ui,jj .

rather than the Helmholtz operator form, m = u − α 2 Div Grad u,

The corresponding Lagrangians are, respectively, 1 lCH (u) = (|u|2 + α 2 (Div u)2 )dxdy. 2

(2.14)

214


and lEPDiff (u) =

1 2

(|u|2 + α 2 | Grad u|2 )dxdy.

(2.15)

This difference was noted in Kruse, Scheurle, and Du [2001], which identified (2.14) as the generalization of (1.4) for water waves in two dimensions. One may also verify this by considering the limit of the Green–Nagdhi equations for small potential energy. (The CH equation arises in this limit. The Lake and Great Lake equations of Camassa, Holm, and Levermore [1996, 1997] also arise in a variant of this limit.) Remarkably, the numerics in Holm and Staley [2003, 2004] show that the solutions for a variety of initial conditions are indistinguishable in these two cases. The initial conditions in Holm and Staley [2003, 2004] were all spatially confined velocity distributions. Notice that this difference affects the choice of Hamiltonian, but the equations are still Euler–Poincaré equations for the diffeomorphism group and the description of the Ansatz (2.8) as a momentum map is independent of this difference in the equations. Figure 2.2 shows the striking reconnection phenomenon seen in the nonlinear interaction between wave-trains, as simulated by numerical solutions of the EPDiff equation and observed for internal waves in the ocean. Figure 2.2(a) shows a frame taken from simulations of the initial value problem for the EPDiff equation in two dimensions, excerpted from Holm and Staley [2003, 2004]. (See also Holm et al. [2003].) Figure 2.2(b) shows the interaction of two internal wave trains propagating at the interface of different density levels in the South China Sea, as observed from the Space Shuttle using synthetic aperture radar, courtesy of A. Liu (2002). Most important, both Figures 2.2(a) and 2.2(b) show nonlinear reconnection occurring in the wave-train interaction as their characteristic feature. Figure 2.3 shows a sequence of snapshots illustrating the reconnection phenomenon for singular solutions of EPDiff in two dimensions.4 Interactions among internal waves are generally thought to be described by the KP equation, and so any relations among the KP equation, the EPDiff equation and the 2D CH equation would be of great interest to explore; see Liu et al. [1998]. The derivations of the KP equation and the CH equation differ in the way the gradients of their transverse motions are treated in the asymptotics—order O() for KP and order O(1) for CH; thus some difference in their solution behavior is to be expected.

3 Smoothness of the Lagrangian equations The one-dimensional case Based on a formal argument given in Holm, Marsden, and Ratiu [1998a], it was shown in Shkoller [1998] that the CH equation (1.2) in Lagrangian variables defines 4 Figures 2.2(a) and 2.3 were kindly supplied by Martin Staley.


(a)

215

(b)

Fig. 2.2. Comparison of evolutionary EPDiff solutions in two dimensions (a) and Synthetic Aperture Radar observations by the Space Shuttle of internal waves in the South China Sea (b). Both figures show nonlinear reconnection occurring in the wave-train interaction as their characteristic feature.

Fig. 2.3. A single collision is shown to produce reconnection as the faster wave front segment initially moving southwest along the diagonal expands, curves and obliquely overtakes the slower one, which was initially moving rightward (east). This reconnection illustrates one of the collision rules for singular solutions of the two-dimensional EPDiff flow. See Holm and Staley [2004] for a complete treatment.

216


a smooth vector field. (That is, one obtains an evolution equation with no derivative loss.) This means one can show using ODE methods that the initial value problem is well posed, and one may also establish other important properties of the equations, provided the data is sufficiently smooth. As above, we write the relation between m and u as m = Qop u, so that in the one-dimensional case, Qop is the operator Qop = Id −α 2 ∂xx . We first recall how the equations are transformed into Lagrangian variables. Introduce the one-parameter curve of diffeomorphisms η(x0 , t) defined implicitly by ∂ η(x0 , t) = u(η(x0 , t), t), ∂t

(3.1)

so that η is a geodesic in the group of diffeomorphisms of R (or, with periodic boundary conditions, of the circle S 1 ) equipped with the right invariant metric equaling the H 1 metric at the identity. We compute the second time derivative of η in a straightforward way by differentiating (3.1) using the chain rule ∂ 2η ∂u . = uux + 2 ∂t ∂t Acting on this equation with Qop and using the definition m = Qop u yields Qop

∂ 2η ∂m = Qop (uux ) − u∂x (Qop u) + umx + ∂t ∂t 2 = [Qop , u∂x ]u − 2mux = −3α 2 ux uxx − 2mux = −α 2 ux uxx − 2uux ,

where the third step uses the commutator relation calculated from the product rule, [Qop , u∂x ]u = −3α 2 ux uxx . Hence, the preceding equation becomes ∂ 2η 1 = − Q−1 ∂x (α 2 u2x + 2u2 ). 2 op ∂t 2

(3.2)

The important point about this equation is that the right-hand side has no derivative loss for α > 0. That is, if u is in the Sobolev space H s for s > 5/2, then the right-hand side is also in the same space. Regarding the right-hand side as a function of η and ∂η/∂t, we see that it is plausible that the second-order evolution equation (3.2) for η defines a smooth ODE on the group of H s diffeomorphisms. (This argument requires the use of, for example, weighted Sobolev spaces in the case x ∈ R.) The above is the essence of the argument given in Shkoller [1998], Remark 3.5, which in turn makes use of the type of arguments found in Ebin and Marsden [1970] for the incompressible case and which shows, by a more careful argument, that the


217

spray is smooth if s > 3/2. However, one should note that the complete argument is not quite so simple (as in the case of incompressible fluids). A subtlety arises because smoothness means as a function of η, η. ˙ Hence, one must express u in terms of η, namely, through the relation ut = η˙ t ◦ ηt−1 , where the subscript t here denotes that this argument is held fixed, and is not a partial derivative. Doing this, one sees that, while there is clearly no derivative loss, the right-hand side of (3.2) does involve ηt−1 and the map ηt → ηt−1 is known to not be smooth. Nevertheless, the combination that appears in (3.2) is, quite remarkably, a smooth function of η, η˙ as is shown by arguments in Ebin and Marsden [1970]. The n-dimensional case The above argument readily generalizes to n-dimensions, which we shall present in the case of Rn or the flat n-torus Tn for simplicity. Namely, we still have the relation ∂ η(x0 , t) = u(η(x0 , t), t), ∂t between η and u. Consequently, we may compute the second partial time derivative of η in the usual fashion using the chain rule ∂u ∂ 2η . = u · ∇u + ∂t ∂t 2 Therefore, as in the one-dimensional case, we get ∂ 2η ∂m . = [Qop , (u · ∇)]u + u · ∇m + 2 ∂t ∂t Calculating the commutator relation in n-dimensions gives Qop

[Qop , (u · ∇)]u = −α 2 div(∇u · ∇u + ∇u · ∇uT ) + α 2 (∇u) · ∇ div u or, in components, ([Qop , (u · ∇)]u)i = −α 2 ∂k (ui,j uj,k + ui,j uk,j ) + α 2 (ui,j )∂j div u,

(3.3)

with a sum on repeated indices. Upon substituting the preceding commutator relation, the EPDiff equation (2.1) and the vector calculus identity 1 2 α2 T 2 T 2 |u| + |∇u| , (3.4) −∇u · m = α div(∇u · ∇u) − ∇ 2 2 then imply the n-dimensional result Qop

∂ 2η ∂t 2

1 T T T 2 = −α div ∇u · ∇u + ∇u · ∇u − ∇u · ∇u − ∇u (div u) + Id |∇u| 2 1 − u(div u) − ∇|u|2 . 2 A similar computation holds on a Riemannian manifold (or in curvilinear coordinates) 2

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in terms of covariant derivatives. This form of the EPDiff equation is useful for interpreting some of its solution behavior. As in the one-dimensional case, the crucial point is that the right-hand side involves at most second derivatives of u; so there is no derivative loss in the expression for ∂ 2 η/∂t 2 . This is the main idea behind the proof of smoothness. The technical details for the n-dimensional case can be provided following the arguments for the one-dimensional or incompressible cases, as indicated above. This leads to the following result. Proposition 3.1. For s > (n/2) + 1, and M a compact Riemannian manifold, the EPDiff equations as second-order equations on the H s -Diff (M) group, define a smooth spray. In particular, this implies the following: 1. The EPDiff equations are locally well posed (for short time) for initial data in H s . 2. Two nearby diffeomorphisms can be joined by a unique curve (lying in the neighborhood of these diffeomorphisms) which is the flow of a solution of the EPDiff equations for time ranging from 0 to 1. 3. With initial data in H s , the solutions of the EPDiff equation are C ∞ in time. For example, if M is the three torus, this corresponds to solutions in R3 with spatially periodic boundary conditions. By using methods such as those of Cantor [1975], we one may reasonably expect to establish a similar result for Rn in weighted (Nirenberg–Walker) Sobolev spaces. While local well posedness of the EPDiff equations is a fairly routine matter from the PDE point of view, the other properties are not so simple to obtain by classical PDE methods. In the sections that follow, we will be interested in nonsmooth data. This is in stark contrast to the preceding discussion, which requires initial data that is at least C 1 . Remarkably, the same smoothness results hold for the case of the LAE-α (Lagrangian averaged Euler) equations, a set of incompressible equations in which small scale fluctuations whose size is of order α are averaged. One can view the LAE-α equations as the incompressible version of the EPDiff equations. This smoothness property for the LAE-α equations was shown by Shkoller [1998] for regions with no boundary and for regions with boundary (for various boundary conditions), it was shown in Marsden et al. [2000]. However, unlike the incompressible case, the results apparently do not hold if α is zero (as was also noted in Shkoller [1998]). This sort of smoothness result also appears not to hold for many other equations, such as the KdV equation, even though it too can be realized as Euler–Poincaré equations on a Lie algebra, or as geodesics on a group, in this case the Bott–Virasoro group, as explained in Marsden and Ratiu [1999] and references therein. Development of singularities The smoothness property just discussed does not preclude the development in finite time of singular solutions from smooth localized initial data, as was indicated in


219

Figure 2.1. To capture the local singularities in the EPDiff solution (either verticality in slope, or discontinuities in its spatial derivative) that develop in finite time from arbitrarily smooth initial conditions, one must enlarge the solution class of interest by considering weak solutions. There are a number of papers on weak solutions of the CH equation (such as, for instance, Xin and Zhang [2000]) which we will not survey here. We just mention that the theory is not yet complete, as it is still unknown in what sense one may define global unique weak solutions to the CH equations in H 1 —only results that have an energy conservation theorem and allow for the head-on collision of two peakons would be considered interesting. As discussed in Alber, Camassa, Fedorov, Holm, and Marsden [2001] for the CH equation, one most likely must consider weak solutions in the spacetime sense. The steepening lemma of Camassa and Holm [1993] proves that in one dimension any initial velocity distribution whose spatial profile has an inflection point with negative slope (for example, any antisymmetric smooth initial distribution of velocity on the real line) will develop a vertical slope in finite time. Note that the peakon solution (2.7) has no inflection points, so it is not subject to the steepening lemma. However, the steepening lemma underlies the mechanism for forming these singular solutions, which are continuous but have discontinuous spatial derivatives; they also lie in H 1 and have finite energy. We conclude that solutions with initial conditions in H s with s > (n/2) + 1 go to infinity in the H s norm in finite time, but remain in H 1 and presumably continue to exist in a weak spacetime sense for all time in H 1 . Numerical evidence in higher dimensions and the inverse scattering solution for the CH equation in one dimension (the latter has only discrete eigenvalues, corresponding to peakons) both suggest that the singular solutions completely dominate the time-asymptotic dynamics of the initial value problem (IVP). This singular IVP behavior is one of the main discoveries of Camassa and Holm [1993]. This singular behavior has drawn a great deal of mathematical interest to the CH equation and its relatives, such as EPDiff. The other properties of CH—its complete integrability, inverse scattering transform, connections to algebraic geometry and elliptical billiards, bi-Hamiltonian structure—are, of course, all interesting too. However, the requirement of dealing with singularity as its main solution phenomenon is the primary aspect of CH (and EPDiff). We aim to show that many of the properties of these singular solutions of CH and EPDiff are captured by recognizing that the singular solution ansatz itself is a momentum map. This momentum map property explains, for example, why the singular solutions (2.8) form an invariant manifold for any value of N and why their dynamics form a Hamiltonian system. In one dimension, the complete integrability of the CH equation as a Hamiltonian system and its soliton paradigm explain the emergence of peakons in the CH dynamics. Namely, their emergence reveals the initial condition’s soliton (peakon) content. However, beyond one dimension, we do not have an explicit mechanism for explaining why only singular solution behavior emerges in numerical simulations. One hopes that eventually a theory will be developed for explaining this observed singular solution phenomenon in higher dimensions. Such a theory might, for example, parallel the well-known explanation of the formation of shocks for hyperbolic

220


partial differential equations. (Note, however, that EPDiff is not hyperbolic, because the relation u = G ∗ m between its velocity and momentum is nonlocal.) In the remainder of this work, we shall focus on the momentum map properties of the invariant manifold of singular solutions (2.8) of the EPDiff equation.

4 Singular solution momentum map The momentum ansatz (2.8) is a momentum map The purpose of this section is to show that the solution ansatz (2.8) for the momentum vector in the EPDiff equation (2.1) defines a momentum map for the action of the group of diffeomorphisms on the support sets of the Dirac delta functions. These support sets are the analogs of points on the real line for the CH equation in one dimension. They are points, curves, or surfaces in Rn for the EPDiff equation in n dimensions. This result, as we shall discuss in greater detail later, shows that the solution ansatz (2.8) fits naturally into the scheme of Clebsch, or canonical variables in the sense advocated by Marsden and Weinstein [1983] as well as showing that these singular solutions evolve on special coadjoint orbits for the diffeomorphism group. One can summarize by saying that the map that implements the canonical (Q, P) variables in terms of singular solutions is a (cotangent bundle) momentum map. Such momentum maps are Poisson maps; so the canonical Hamiltonian nature of the dynamical equations for (Q, P) fits into a general theory which also provides a framework for suggesting other avenues of investigation. Theorem 4.1. The momentum ansatz (2.8) for measure-valued solutions of the EPDiff equation (2.1), defines an equivariant momentum map JSing : T ∗ Emb(S, Rn ) → X(Rn )∗ that we will call the singular solution momentum map. We shall explain the notation used in this statement in the course of the proof. Right away, however, we note that the sense of “defines’’ is quite simple, namely, expressing m in terms of Q, P (which are, in turn, functions of s) can be regarded as a map from the space of (Q(s), P(s)) to the space of m’s. We shall give two proofs of this result from two rather different points of view. The first proof below uses the formula for a momentum map for a cotangent lifted action, while the second focuses on a Poisson bracket computation. Each proof also explains the context in which one has a momentum map. (See Marsden and Ratiu [1999] for general background on momentum maps.) First proof . For simplicity and without loss of generality, let us take N = 1 and so suppress the index a. That is, we shall take the case of an isolated singular solution. As the proof will show, this is not a real restriction.


221

To set the notation, fix a k-dimensional manifold S with a given volume element and whose points are denoted s ∈ S. Let Emb(S, Rn ) denote the set of smooth embeddings Q : S → Rn . (If the EPDiff equations are taken on a manifold M, replace Rn with M.) Under appropriate technical conditions, which we shall just treat formally here, Emb(S, Rn ) is a smooth manifold. (See, for example, Ebin and Marsden [1970] and Marsden and Hughes [1983] for a discussion and references.) The tangent space TQ Emb(S, Rn ) to Emb(S, Rn ) at the point Q ∈ Emb(S, Rn ) is given by the space of material velocity fields, namely, the linear space of maps V : S → Rn that are vector fields over the map Q. The dual space to this space will be identified with the space of one-form densities over Q, which we shall regard as maps P : S → (Rn )∗ . In summary, the cotangent bundle T ∗ Emb(S, Rn ) is identified with the space of pairs of maps (Q, P). These give us the domain space for the singular solution momentum map. Now we consider the action of the symmetry group. Consider the group G = Diff of diffeomorphisms of the space M in which the EPDiff equations are operating, concretely in our case Rn . Let it act on M by composition on the left. Namely, for η ∈ Diff (Rn ), we let η · Q = η ◦ Q. (4.1) Now lift this action to the cotangent bundle T ∗ Emb(S, Rn ) in the standard way (see, for instance, Marsden and Ratiu [1999] for this construction). This lifted action is a symplectic (and hence Poisson) action and has an equivariant momentum map. We claim that this momentum map is precisely given by the ansatz (2.8). To see this, we will recall and then apply the general formula for the momentum map associated with an action of a general Lie group G on a configuration manifold Q and cotangent lifted to T ∗ Q. First, let us recall the general formula. Namely, the momentum map is the map J : T ∗ Q → g∗ (g∗ denotes the dual of the Lie algebra g of G) defined by J(αq ) · ξ = αq , ξQ (q),

(4.2)

where αq ∈ Tq∗ Q and ξ ∈ g, where ξQ is the infinitesimal generator of the action of G on Q associated to the Lie algebra element ξ , and where αq , ξQ (q) is the natural pairing of an element of Tq∗ Q with an element of Tq Q. Now we apply formula (4.2) to the special case in which the group G is the diffeomorphism group Diff (Rn ), the manifold Q is Emb(S, Rn ) and where the action of the group on Emb(S, Rn ) is given by (4.1). The sense in which the Lie algebra of G = Diff is the space g = X of vector fields is well understood. Hence, its dual is naturally regarded as the space of one-form densities. The momentum map is thus a map J : T ∗ Emb(S, Rn ) → X∗ . To calculate J given by (4.2), we first work out the infinitesimal generators. Let X ∈ X be a Lie algebra element. By differentiating the action (4.1) with respect to η in the direction of X at the identity element we find that the infinitesimal generator is given by XEmb(S,Rn ) (Q) = X ◦ Q. Thus, taking αq to be the cotangent vector (Q, P), equation (4.2) gives

222


J(Q, P), X = (Q, P), X ◦ Q = Pi (s)X i (Q(s))d k s. S

On the other hand, note that the right-hand side of (2.8) (again with the index a suppressed, and with t suppressed as well), when paired with the Lie algebra element X is P(s)δ(x − Q(s))d k s, X = (Pi (s)δ(x − Q(s))d k s)X i (x)d n x n S R S = Pi (s)X i (Q(s)d k s. S

This shows that the expression given by (2.8) is equal to J and so the result is proved.

Second proof . As is standard (see, for example, Marsden and Ratiu [1999]), one can characterize momentum maps by means of the following relation, required to hold for all functions F on T ∗ Emb(S, Rn ), that is, functions of Q and P: {F, J, ξ } = ξP [F ].

(4.3)

In our case, we shall take J to be given by the solution ansatz and verify that it satisfies this relation. To do so, let ξ ∈ X so that the left side of (4.3) becomes 4 5 δF i δF δ i F, Pi (s)ξ i (Q(s))d k s = ξ (Q(s)) − P (s) ξ (Q(s)) d k s. i i δPj δQj S S δQ On the other hand, one can directly compute from the definitions that the infinitesimal generator of the action on the space T ∗ Emb(S, Rn ) corresponding to the vector field ∂ ξ i (x) ∂Q i (a Lie algebra element), is given by (see Marsden and Ratiu [1999], formula (12.1.14)): ∂ i ξ (Q(s)), δQ = ξ ◦ Q, δP = −Pi (s) ∂Q which verifies that (4.3) holds. An important element left out in this proof so far is that it does not make clear that the momentum map is equivariant, a condition needed for the momentum map to be Poisson. The first proof took care of this automatically since momentum maps for cotangent lifted actions are always equivariant and hence Poisson. Thus, to complete the second proof, we need to check directly that the momentum map is equivariant. Actually, we shall only check that it is infinitesimally invariant by showing that it is a Poisson map from T ∗ Emb(S, Rn ) to the space of m’s (the dual of the Lie algebra of X) with its Lie–Poisson bracket. This sort of approach to characterize equivariant momentum maps is discussed in an interesting way in Weinstein [2002]. The following computation accomplishes this methodology by showing directly that the singular solution momentum map is Poisson. To do this we use the canonical


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Poisson brackets for {P}, {Q} and apply the chain rule to compute {mi (x), mj (y)}. Using the notation δk (y) ≡ ∂δ(y)/∂y k , we get {mi (x), mj (y)} +N 3 N a a b b = dsPi (s, t)δ(x − Q (s, t)), ds Pj (s , t)δ(y − Q (s , t)) a=1

=

N

b=1

dsds {Pia (s), Pjb (s )}δ(x − Qa (s))δ(y − Qb (s ))

a,b=1

− {Pia (s), Qbk (s )}Pjb (s )δ(x − Qa (s))δk (y − Qb (s )) − {Qak (s), Pjb (s )}Pia (s)δk (x − Qa (s))δ(y − Qb (s ))

+ {Qak (s), Qb (s )}Pia (s)Pjb (s )δk (x − Qa (s))δ (y − Qb (s )) .

Substituting the canonical Poisson bracket relations {Pia (s), Pjb (s )} = 0, {Qak (s), Qb (s )} = 0, and {Qak (s), Pjb (s )} = δ ab δkj δ(s − s ) into the preceding computation yields {mi (x), mj (y)} +N 3 N = dsPia (s, t)δ(x − Qa (s, t)), ds Pjb (s , t)δ(y − Qb (s , t)) a=1

=

N

b=1

dsPja (s)δ(x − Qa (s))δi (y − Qa (s))

a=1

−

N

dsPia (s)δj (x − Qa (s))δ(y − Qa (s))

a=1

∂ ∂ = − mj (x) i + j mi (x) δ(x − y). ∂x ∂x ∂ ∂ {mi (x), mj (y)} = − mj (x) i + j mi (x) δ(x − y), ∂x ∂x which is readily checked to be the Lie–Poisson bracket on the space of m’s. This completes the second proof of theorem.

Thus

Each of these proofs has shown the following basic fact. Corollary 4.2. The singular solution momentum map defined by the singular solution ansatz, namely,

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JSing : T ∗ Emb(S, Rn ) → X(Rn )∗ is a Poisson map from the canonical Poisson structure on T ∗ Emb(S, Rn ) to the Lie–Poisson structure on X(Rn )∗ . This is perhaps the most basic property of the singular solution momentum map. Some of its more sophisticated properties are outlined in the following section. Pulling back the equations Since the solution ansatz (2.8) has been shown in the preceding corollary to be a Poisson map, the pullback of the Hamiltonian from X∗ to T ∗ Emb(S, Rn ) gives equations of motion on the latter space that project to the equations on X∗ . Thus the basic fact that the momentum map JSing is Poisson explains why the functions Qa (s, t) and Pa (s, t) satisfy canonical Hamiltonian equations. Note that the coordinate s ∈ Rk that labels these functions is a “Lagrangian coordinate’’ in the sense that it does not evolve in time but rather labels the solution. In terms of the pairing ·, · : g∗ × g → R, (4.4) between the Lie algebra g (vector fields in Rn ) and its dual g∗ (one-form densities in Rn ), the following relation holds for measure-valued solutions under the momentum map (2.8), m, u = m · ud n x, L2 pairing for m and u ∈ Rn , =

N

(Pa (s, t) · Pb (s , t))G(Qa (s, t) − Qb (s , t))dsds

a,b=1

=

N

Pa (s, t) ·

a=1

˙ ≡ P, Q,

∂Qa (s, t) ds ∂t (4.5)

˙ ∈ which is the natural pairing between the points (Q, P) ∈ T ∗ Emb(S, Rn ) and (Q, Q) T Emb(S, Rn ). The pullback of the Hamiltonian H [m] defined on the dual of the Lie algebra g∗ , to T ∗ Emb(S, Rn ) is easily seen to be consistent with what we had before: 1 1 m, G ∗ m = P, G ∗ P ≡ HN [P, Q]. (4.6) 2 2 In summary, in concert with the Poisson nature of the singular solution momentum map, we see that the singular solutions in terms of Q and P satisfy Hamiltonian equations and also define an invariant solution set for the EPDiff equations. In fact, H [m] ≡

this invariant solution set is a special coadjoint orbit for the diffeomorphism group, as we shall discuss in the next section.


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Remark. It would be extremely interesting if the smoothness properties explored in Section 3 were also valid on the space T ∗ Emb(S, Rn ). This is obviously valid for the CH equation.

5 Geometry of the momentum map In this section we explore the geometry of the singular solution momentum map discussed in Section 4 in a little more detail. The approach may be stated as follows: simply apply all of the ideas given in Marsden and Weinstein [1983] in a systematic way to the current setting. As in that paper, the treatment is formal, in the sense that there are a number of technical issues in the infinite-dimensional case that are left open. We will mention a few of these as we proceed. Coadjoint orbits We claim that the image of the singular solution momentum map is a coadjoint orbit in X∗ . This means that (modulo some issues of connectedness and smoothness, which we do not consider here) the solution ansatz given by (2.8) defines a coadjoint orbit in the space of all one-form densities, regarded as the dual of the Lie algebra of the diffeomorphism group. These coadjoint orbits should be thought of as singular orbits—that is, due to their special nature, they are not generic. Recognizing them as coadjoint orbits is one way of gaining further insight into why the singular solutions form dynamically invariant sets—it is a general fact that coadjoint orbits in g∗ are symplectic submanifolds of the Lie–Poisson manifold g∗ (in our case X(Rn )∗ ) and, correspondingly, are dynamically invariant for any Hamiltonian system on g∗ . The idea of the proof of our claim is simply this: whenever one has an equivariant momentum map J : P → g∗ for the action of a group G on a symplectic or Poisson manifold P , and that action is transitive, then the image of J is an orbit (or at least a piece of an orbit). This general result, due to Kostant, is stated more precisely in Marsden and Ratiu [1999], Theorem 14.4.5. Roughly speaking, the reason that transitivity holds in our case is because one can “move the images of the manifolds S around at will with arbitrary velocity fields’’ using diffeomorphisms of Rn . Symplectic structure on orbits Recall (from, for example, Marsden and Ratiu [1999]), the general formula for the symplectic structure on coadjoint orbits:

µ (ξg∗ (µ), ηg∗ (µ)) = µ, [ξ, η],

(5.1)

where µ ∈ g∗ is a chosen point on an orbit and where ξ, η are elements of g. We use a plus sign in this formula since we are dealing with orbits for the right action.

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As in Marsden and Weinstein [1983], this line of investigation leads to an explicit formula for the coadjoint orbit symplectic structure in the case of Diff . In the present case, it is a particularly simple and transparent formula. Recall that in the case of incompressible fluid mechanics, this procedure leads naturally to the symplectic (and Poisson) structure for many interesting singular coadjoint orbits, such as point vortices in the plane, vortex patches, vortex blobs (closely related to the planar LAE-α equations) and vortex filaments. An important point is that this structure is independent of how these solutions are parametrized. For the case of the diffeomorphism group, let Om denote the coadjoint orbit through the point m ∈ X∗ (Rn ). Theorem 5.1. The symplectic structure m on Tm Om is given by

m (£u1 m, £u2 m) = − m, [u1 , u2 ]d n x. Proof. We substitute into the general Kirillov–Kostant–Souriau formula (5.1) for the symplectic structure on coadjoint orbits. (As noted above, there is a + sign, since we are dealing with a right invariant system). The only thing needing explanation is that our Lie algebra convention always uses the left Lie bracket. For Diff , this is the negative of the usual Lie bracket, as explained in Marsden and Ratiu [1999].

The momentum map JS and the Kelvin circulation theorem The momentum map JSing involves Diff (Rn ), the left action of the diffeomorphism group on the space of embeddings Emb(S, Rn ) by smooth maps of the target space Rn , namely, Diff (Rn ) : Q · η = η ◦ Q, (5.2) where we recall that Q : S → Rn . As above, the cotangent bundle T ∗ Emb(S, Rn ) is identified with the space of pairs of maps (Q, P), with Q : S → Rn and P : S → T ∗ Rn . However, there is another momentum map JS associated with the right action of the diffeomorphism group of S on the embeddings Emb(S, Rn ) by smooth maps of the “Lagrangian labels’’ S (fluid particle relabeling by η : S → S). This action is given by Diff (S) : Q · η = Q ◦ η. (5.3) The infinitesimal generator of this right action is d XEmb(S,Rn ) (Q) = Q ◦ ηt = T Q ◦ X, dt t=0

(5.4)

where X ∈ X is tangent to the curve ηt at t = 0. Thus, again taking N = 1 (so we suppress the index a) and also letting αq in the momentum map formula (4.2) be the cotangent vector (Q, P), one computes JS : JS (Q, P), X = (Q, P), T Q · X


=

Pi (s) S

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∂Qi (s) m X (s)d k s ∂s m

=

X(P(s) · dQ(s))d k s k P(s) · dQ(s) ⊗ d s, X(s) = S

S

= P · dQ, X. Consequently, the momentum map formula (4.2) yields JS (Q, P) = P · dQ,

(5.5)

with the indicated pairing of the one-form density P · dQ with the vector field X. We have set things up so that the following is true. Proposition 5.2. The momentum map JS is preserved by the evolution equations (2.12) for Q and P. Proof. It is enough to notice that the Hamiltonian HN in equation (2.13) is invariant under the cotangent lift of the action of Diff (S); it merely amounts to the invariance of the integral over S under reparametrization, that is, the change of variables formula; keep in mind that P includes a density factor.

This result is similar to the Kelvin–Noether theorem for circulation of an ideal 2 fluid, which may be written as = c(s) D(s)−1 P(s) · dQ(s) for each Lagrangian circuit c(s), where D is the mass density and P is again the canonical momentum density. This similarity should come as no surprise, because the Kelvin–Noether theorem for ideal fluids arises from invariance of Hamilton’s principle under fluid parcel relabeling by the same right action of the diffeomorphism group, as in (5.3). Note that, being an equivariant momentum map, the map JS , as with JSing , is also a Poisson map. That is, substituting the canonical Poisson bracket into relation (5.5); that is, the relation M(x) = i Pi (x)∇Qi (x) yields the Lie–Poisson bracket on the space of M’s. We use the different notations m and M because these quantitites are analogous to the body and spatial angular momentum for rigid body mechanics. In fact, the quantity m is given by the solution Ansatz; specifically, m = JSing (Q, P) gives the singular solutions of the EPDiff equations, while M(x) = JS (Q, P) = i i Pi (x)∇Q (x) is a conserved quantity. In the language of fluid mechanics, the expression of m in terms of (Q, P) is an example of a “Clebsch representation,’’ which expresses the solution of the EPDiff equations in terms of canonical variables that evolve by standard canonical Hamilton equations. This has been known in the case of fluid mechanics for more than 100 years. For modern discussions of the Clebsch representation for ideal fluids, see, for example, Holm and Kupershmidt [1983]; Marsden and Weinstein [1983]. One more remark is in order, namely, that the special case in which S = M is of course allowed. In this case, Q corresponds to the map η itself and P just corresponds to its conjugate momentum. The quantity m corresponds to the spatial

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(dynamic) momentum density (that is, right translation of P to the identity), while M corresponds to the conserved “body’’ momentum density (that is, left translation of P to the identity). Dual pairs For reasons that are similar to those for incompressible fluids presented in Marsden and Weinstein [1983], the singular solution momentum map JSing : T ∗ Emb(S, Rn ) → X(Rn )∗ forms one leg of a formal dual pair. We use the words formal dual pair since, in the infinite-dimensional case, the proper mathematical underpinnings for the theory of dual pairs has not yet been developed. Even in the finite-dimensional case, there are nontrivial issues to be aware of since dual pairs were studied in the basic paper of Weinstein [1983b]; we refer to Ortega and Ratiu [2004], Chapter 11, as well as Blaom [2001] and Ortega [2003] for background, references and a summary of the current state-of-the-art in this topic. These works show the subtlety of the dual pairs notion, even in finite dimensions, let alone for the infinite-dimensional problem we are dealing with here. The point is that, as we have seen, there is another group that acts on Emb(S, Rn ), namely, the group Diff (S) of diffeomorphisms of S, which acts on the right, while Diff (Rn ) acted by composition on the left (and this gave rise to our singular solution momentum map JSing ). As explained above, the action of Diff (S) from the right gives us the momentum map JS : T ∗ Emb(S, Rn ) → X(S)∗ . We now assemble both momentum maps into one figure as follows: T ∗ Emb(S, M) JSing X(M)∗

@

@ JS @ R @ X(S)∗

These maps have the formal dual pair property, namely, that the kernel of the derivatives of each map at a given point are symplectic orthogonals of one another (see Weinstein [1983a]). Sometimes, as in Ortega and Ratiu [2004], this is called the Lie–Weinstein property. Formal proof of the dual pair property. The reduction lemma of Marsden and Weinstein [1974] states that the kernel of the derivative of a momentum map is the symplectic orthogonal of the group orbit. As a consequence, if the group associated to each leg of a potential dual pair of momentum maps acts transitively on the level set of its partner momentum map, then one has a dual pair. In our case, fixing JS at a value, say M, means, according to equation (5.5), that we fix the value of P · dQ. However, as we already noted above, the group Diff (M) acts transitively on the space of Q’s because one can “move the singular surfaces around at will’’ by means of diffeomorphisms of M. The constraint of fixing P · dQ is exactly what


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one needs to transform the P’s properly by means of the cotangent lift (recall that cotangent lift actions are characterized by preserving the canonical one-form). Thus, at least formally, Diff (M) acts transitively on level sets of JS . Similarly, one sees that Diff (S) acts transitively on level sets of JSing since fixing JSing corresponds to fixing the image surface, leaving one only with the parametrization freedom, so that Diff (S) acts transitively on that set.

This is a marvelous framework; it clarifies, among other things, the fact that the parameterization of the singular solutions m in terms of Q and P are Clebsch variables in the sense given in Marsden and Weinstein [1983] and that the diffeomorphism group of S corresponds to the gauge group of that Clebsch representation. Also, notice that when we write the singular solutions in Q-P space, we are finding solutions that are collective and so all the properties of collectivization are valid. See Marsden and Ratiu [1999] for a general discussion and references to the original work of Guillemin and Sternberg on this topic. As explained in Marsden and Weinstein [1983], reduction by the group associated with one leg in a dual pair corresponds to coadjoint orbits on the other leg. Thus the momentum map JS captures the analog of the Kelvin circulation theorem of fluid mechanics, as well as its singular version. It would be interesting to explore in more detail this singular analog of the Kelvin circulation theorem for fluids. The ideal fluid dual pair In Marsden and Weinstein [1983] a dual pair was investigated that captures certain singular situations in fluid mechanics, such as the motion of point vortices in the plane. The general dual pair that generalizes that planar case is the following: Emb(S, P ) @

JP X(P )∗sym

@ JS @ R @ X(S)∗div

Here, S is a volume manifold , that is a manifold with a volume element, while P is a symplectic manifold . The map JP is the momentum map for the left action of the group of symplectic diffeomorphisms on P , while JS is the momentum map for the right action of the group of volume-preserving diffeomorphisms. This is a very beautiful dual pair, but is not the same, of course, as the dual pair we found above. In our case, P = T ∗ M was a cotangent bundle and we identified Emb(S, P ) with T ∗ Emb(S, M). Also, we always dealt with symplectic diffeomorphisms that were cotangent lifts, while in the above dual pair of Marsden and Weinstein [1983], they are general symplectic diffeomorphisms.

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Relation with ideas of Donaldson Whereas Marsden and Weinstein [1983] focused on ideas related to the dual pair picture, the leg in the above diagram given by the map JS is discussed from various interesting viewpoints in Donaldson [1999]. In particular, that work (apparently being unaware of the above dual pair of Marsden and Weinstein [1983]) makes a number of intriguing comments, including noting that nontrivial topology can cause the momentum map JS to be nonequivariant (so there are links with the Calabi theory). Donaldson also studies reduction and makes links with Kähler geometry, hyper-Kähler geometry, double bracket gradient flows, mean curvature flows, and other intriguing topics. As pointed out by Tony Bloch, there are also interesting links of Donaldson’s paper with the Toda flow and factorization problems. We believe that the pursuit of further connections within the circle of ideas for momentum maps should be a source of inspiration for new research in the context of this paper. For example, this pursuit may lead to new insight into the integrability of the dynamical systems governing these singular solutions. It seems that we are looking at the tip of a rather large and beautiful iceberg.

6 Challenges, future directions, and speculations Numerical issues: Geometric integrators The computations of Martin Staley that illustrated several points in this paper are discussed in detail by Holm and Staley [2003, 2004]. These computations make use of both mimetic differencing and reversibility in a critical way, and this is important for accurate numerical simulations. In other words, integrators that respect the basic geometry underlying the problem obtained accurate singular solutions in numerical simulations. It would be interesting to pursue this aspect further and also incorporate discrete exterior calculus and variational multisymplectic integration methods (see Desbrun et al. [2003] as well as Marsden et al. [1998] and Lew et al. [2003]). Analytical issues: Geodesic incompleteness of H 1 EPDiff The emergence in finite time of singular solutions from smooth initial data observed numerically in Holm and Staley [2003, 2004] indicates that the diffeomorphism group with respect to the right invariant H 1 metric is geodesically incomplete when the diffeomorphism group has the H s topology s > (n/2) + 1. The degree of its geodesic incompleteness is not known, but we suspect that almost all EPDiff geodesics in H 1 cannot be extended indefinitely. This certainly holds in one spatial dimension, where the discreteness of the CH isospectrum implies that asymptotically in time the CH solution arising from any confined smooth initial velocity data consists only of peakons. It is an important challenge to find a context in which one can put the H 1 topology on the diffeomorphism group and reestablish geodesic completeness. The numerics suggests that this might be possible, while known existence theorems, even for the CH equation are not yet capable of showing this—to the best of our knowledge.


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Reversible reconnections of the singular EPDiff solutions EPDiff is a reversible equation, and the collisions of its peakon solutions on the line R1 (or the circle S 1 ) are known to be reversible. The reconnections of the singular EPDiff solutions observed numerically in Holm and Staley [2003, 2004] in periodic domains T2 and T3 are also reversible, and this was used as a test of the numerical method. Reversibility of its reconnections distinguishes the singular solutions of EPDiff from vortex fluid solutions and shocks in fluids, whose reconnections apparently require dissipation, and so are not reversible. The mimetic finite differencing scheme used for the numerical computation of EPDiff solutions in Holm and Staley [2003, 2004] was indeed found to be reversible for overtaking collisions, but it was found to be only approximately reversible for head-on collisions, which are much more challenging for numerical integration schemes. Applications of EPDiff singular solutions in image processing The singular EPDiff solutions correspond to outlines (or cartoons) of images in applications of geodesic flow for the template, or pattern matching approach. The dynamics of the singular EPDiff solutions described by the momentum map (2.8) introduces the paradigm of momentum exchange in soliton collisions into the mechanics and analysis of image processing by template matching. (See Holm, Trouvé, Ratnanather, and Younes [2004] for more discussions of this new paradigm for image processing.) First, the momentum representation of the image outlines is nonredundant. That is, the momentum has exactly the same dimension as the matched structures; so there is no redundancy of the representation. Second, the reversibility of the collisions among singular solutions and their reconnections under EPDiff flow assures the preservation of the information contained in the image outlines. In addition, the invariance of the manifold of N singular solutions under EPDiff assures that the fidelity of the image is preserved in the sense of approximation theory. That is, an N soliton approximation of the image outlines remains so, throughout the EPDiff flow. A natural approach for numerically simulating EPDiff flows in image processing is to use multisymplectic algorithms. The preservation of the space–time multisymplectic form by these algorithms introduces an initial-value, final-value formulation of the numerical solution procedure that is natural for template matching. Rigorous Poisson structures In Vasylkevych and Marsden [2003], the question of the (rigorous) Poisson nature of the time t map of the flow of the Euler equations for an ideal fluid in appropriate Sobolev spaces is explored. Given the smoothness properties in Section 3, it seems reasonable that similar properties should also hold for the EPDiff equations. However, as mentioned earlier, these smoothness properties do not preclude the emergence of singular solutions from smooth initial data in finite time, because of the possibility for geodesic incompleteness.

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Other groups The general setting of this paper suggests that perhaps one should look for similar measure-valued or singular solutions associated with other problems, including geodesic flows on the group of symplectic diffeomorphisms (relevant for plasma physics, as in Marsden and Weinstein [1982]), Bott–Virasoro central extensions and supersymmetry groups. Scattering It might be interesting to explore the relation of the singular solution momentum map (2.8) to integrability and scattering data. For example, see Vaninsky [2003] for an interesting discussion of the Poisson bracket for the scattering data of CH in 1D. This turns out to be the Atiyah–Hitchin bracket, which is also related to the Toda lattice, and this fascinating observation leads to an infinite-dimensional version of Jacobi elliptic coordinates. Other issues Of course, there are many other issues remaining to explore that are suggested by the above setting, such as convexity of the momentum map, its extension to Riemannian manifolds, and so on. We shall, however, leave these issues for other publications and other researchers. Acknowledgments We are very grateful to Alan Weinstein for his collaboration, help and inspiring discussions over the years. We thank Martin Staley for letting us illustrate some important points using his computations. We also thank Anthony Bloch, Simon Donaldson, Jonathan Munn, Tudor Ratiu, and Richard Thomas for valuable advice and comments.

References M. Alber, R. Camassa, Y. Fedorov, D. Holm, and J. E. Marsden [2001], The complex geometry of weak piecewise smooth solutions of integrable nonlinear PDE’s of shallow water and Dym type, Comm. Math. Phys., 221, 197–227. M. S. Alber and J. E. Marsden [1992], On geometric phases for soliton equations, Comm. Math. Phys., 149, 217–240. V. I. Arnold [1966], Sur la géométrie différentielle des groupes de Lie de dimenson infinie et ses applications à l’hydrodynamique des fluids parfaits, Ann. Inst. Fourier Grenoble, 16, 319–361. A. D. Blaom [2001], A Geometric Setting for Hamiltonian Perturbation Theory, Memoirs of the American Mathematical Society, Vol. 727, Americal Mathematical Society, Providence, RI. R. Camassa and D. D. Holm [1993],An integrable shallow water equation with peaked solitons, Phys. Rev. Lett., 71, 1661–1664.


233

R. Camassa, D. D. Holm and J. M. Hyman [1994], A new integrable shallow water equation, Adv. Appl. Mech., 31, 1–33. R. Camassa, D. D. Holm, and C. D. Levermore [1996], Long-time effects of bottom topography in shallow water, Phys. D, 98, 258–286. R. Camassa, D. D. Holm, and C. D. Levermore [1997], Long-time shallow-water equations with a varying bottom, J. Fluid Mech., 349, 173–189. M. Cantor [1975], Perfect fluid flows over R n with asymptotic conditions, J. Functional Anal., 18, 73–84. T. Courant and A. Weinstein [1988], Beyond Poisson structures, in Action hamiltoniennes de groupes: Troisième théorème de Lie (Lyon, 1986), Travaux en Cours, Vol. 27, Hermann, Paris, 39–49. M. Desbrun, A. N. Hirani, M. Leok, and J. E. Marsden [2003], Discrete Exterior Calculus, preprint. S. K. Donaldson [1999], Moment maps and diffeomorphisms, Asian J. Math., 3, 1–15. H. R. Dullin, G. A. Gottwald, and D. D. Holm [2001], An integrable shallow water equation with linear and nonlinear dispersion, Phys. Rev. Lett., 87, 194501–194504. H. R. Dullin, G. A. Gottwald, and D. D. Holm [2003], Camassa–Holm, Korteweg– de Vries-5 and other asymptotically equivalent equations for shallow water waves, Fluid Dynam. Res., 33, 73–95. H. R. Dullin, G. A. Gottwald, and D. D. Holm [2004], On asymptotically equivalent shallow water wave equations, Phys. D, 190, 1–14. D. G. Ebin and J. E. Marsden [1970], Groups of diffeomorphisms and the motion of an incompressible fluid, Ann. Math., 92, 102–163. O. Fringer and D. D. Holm [2001], Integrable vs. nonintegrable geodesic soliton behavior, Phys. D, 150, 237–263. A. Hirani, J. E. Marsden, and J. Arvo [2001], Averaged Template Matching Equations, Lecture Notes in Computer Science, Vol. 2134, Springer-Verlag, New York, 528– 543. D. D. Holm and B. A. Kupershmidt [1983], Poisson brackets and Clebsch representations for magnetohydrodynamics, multifluid plasmas, and elasticity, Phys. D, 6, 347–363. D. D. Holm, J. E. Marsden, and T. S. Ratiu [1998a], The Euler–Poincaré equations and semidirect products with applications to continuum theories, Adv. Math., 137, 1–81. D. D. Holm, J. E. Marsden and T. S. Ratiu [1998b], Euler–Poincaré models of ideal fluids with nonlinear dispersion, Phys. Rev. Lett., 349, 4173–4177. D. D. Holm, J. E. Marsden, and T. S. Ratiu [2002], The Euler–Poincaré equations in geophysical fluid dynamics, in J. Norbury and I. Roulstone, eds., Large-Scale Atmosphere-Ocean Dynamics II: Geometric Methods and Models, Cambridge University Press, Cambridge, UK, 251–300. D. D. Holm, J. E. Marsden, T. S. Ratiu, and A. Weinstein [1985], Nonlinear stability of fluid and plasma equilibria, Phys. Rep., 123, 1–196. D. D. Holm, V. Putkaradze, and S. N. Stechmann [2003], Rotating concentric circular peakons, Nonlinearity, submitted; http://arxiv.org/abs/nlin.SI/0312012/9801015.

234


D. D. Holm, J. T. Ratnanather, A. Trouvé, and L. Younes [2004], Solitons in computational anatomy, NeuroImage, to appear. D. D. Holm and M. F. Staley [2003], Wave structures and nonlinear balances in a family of evolutionary PDEs, SIAM J. Appl. Dynam. Systems, 2, 323–380. D. D. Holm and M. F. Staley [2004], Momentum dynamics of filaments and surfaces in a set of 2 + 1 and 3 + 1 evolutionary PDEs, in preparation. Y. Kodama [1985], On integrable systems with higher order corrections, Phys. Lett. A, 107, 245–249. Y. Kodama [1985a], Normal forms for weakly dispersive wave equations, Phys. Lett. A, 112, 193–196. Y. Kodama [1987], On solitary-wave interaction, Phys. Lett. A, 123, 276–282. H. P. Kruse, J. Scheurle, and W. Du [2001], A two-dimensional version of the CH equation, in D. Bambusi, G. Gaeta, and M. Cadoni, eds., Symmetry and Perturbation Theory: SPT 2001, World Scientific, New York, 120–127. A. Lew, J. E. Marsden, M. Ortiz, and M. West [2003], Asynchronous variational integrators, Arch. Rational Mech. Anal., 167, 85–146. A. K. Liu, Y. S. Chang, M. K. Hsu, and N. K. Liang [1998], Evolution of nonlinear internal waves in East and South China Seas, J. Geophys. Res., 103, 7995–8008. J. E. Marsden and T. J. R. Hughes [1983], Mathematical Foundations of Elasticity, Prentice–Hall, Engelwood Cliffs, NJ; reprinted by Dover Publications, New York, 1994. J. E. Marsden, G. W. Patrick, and S. Shkoller [1998], Multisymplectic geometry, variational integrators and nonlinear PDEs, Comm. Math. Phys., 199, 351–395. J. E. Marsden and T. S. Ratiu [1999], Introduction to Mechanics and Symmetry, 2nd ed., Texts in Applied Mathematics, Vol. 17, Springer-Verlag, New York; 1st ed., 1994. J. E. Marsden, T. Ratiu, and S. Shkoller [2000], The geometry and analysis of the averaged Euler equations and a new diffeomorphism group, Geom. Functional Anal., 10, 582–599. J. E. Marsden, T. S. Ratiu, and A. Weinstein [1984], Semi-direct products and reduction in mechanics, Trans. Amer. Math. Soc., 281, 147–177. J. E. Marsden and A. Weinstein [1974], Reduction of symplectic manifolds with symmetry, Rep. Math. Phys., 5, 121–130. J. E. Marsden and A. Weinstein [1982], The Hamiltonian structure of the Maxwell– Vlasov equations, Phys. D, 4, 394–406. J. E. Marsden and A. Weinstein [1983], Coadjoint orbits, vortices and Clebsch variables for incompressible fluids, Phys. D, 7, 305–323. M. I. Miller, A. Trouvé, and L. Younes [2002], On the metrics and Euler-Lagrange equations of computational anatomy, Ann. Rev. Biomed. Engrg., 4, 375–405. D. Mumford [1998], Pattern theory and vision, in Questions mathématiques en traitement du signal et de l’image, Institut Henri Poincaré, Paris, Chapter 3, 7–13. J.-P. Ortega [2003], Singular dual pairs, Differential Geom. Appl., 19, 61–95. J.-P. Ortega and T. S. Ratiu [2004], Momentum Maps and Hamiltonian Reduction, Progress in Mathematics, Vol. 232, Birkhäuser, Boston.


235

S. Shkoller [1998], Geometry and curvature of diffeomorphism groups with H 1 metric and mean hydrodynamics, J. Functional Anal., 160, 337–365. K. L. Vaninsky [2002], TheAtiyah–Hitchin bracket and the open Toda lattice, J. Geom. Phys., 46-3 (2003), 283–307. K. L. Vaninsky [2003], The Camassa–Holm equation on the line and Jacobi elliptic coordinates, preprint, 2003; ArXiv:math-ph/0303063. S. Vasylkevych and J. E. Marsden [2003], The Lie–Poisson structure of the Euler equations of an ideal fluid, preprint. A. Weinstein [1971], Symplectic manifolds and their Lagrangian submanifolds, Adv. Math., 6, 329–346; see also Bull. Amer. Math. Soc., 75 (1969), 1040–1041. A. Weinstein [1973], Normal modes for nonlinear Hamiltonian systems, Invent. Math., 20, 47–57. A. Weinstein [1977], Lectures on Cymplectic Manifolds, CBMS Regional Conference Series in Mathematics, Vol. 29, Conference Board of the Mathematical Sciences, Washington, DC. A. Weinstein [1978], Bifurcations and Hamilton’s principle, Math. Z., 159, 235–248. A. Weinstein [1983a], Sophus Lie and symplectic geometry, Expo. Math., 1, 95–96. A. Weinstein [1983b], The local structure of Poisson manifolds, J. Differential Geom., 18, 523–557. A. Weinstein [1984], Stability of Poisson–Hamilton equilibria, Contemp. Math., 28, 3–14. A. Weinstein [1990], Connections of Berry and Hannay type for moving Lagrangian submanifolds, Adv. Math., 82, 133–159. A. Weinstein [1996], Lagrangian mechanics and groupoids, Fields Inst. Comm., 7, 207–231. A. Weinstein [2002], Geometry of Momentum, preprint; ArXiv:math/ SG0208108 v1. Z. Xin and P. Zhang [2000], On the weak solutions to a shallow water equation, Comm. Pure Appl. Math., 53, 1411–1433.

Higher homotopies and Maurer–Cartan algebras: Quasi-Lie–Rinehart, Gerstenhaber, and Batalin–Vilkovisky algebras Johannes Huebschmann Université des Sciences et Technologies de Lille UFR de Mathématiques, CNRS-UMR 8524 F-59 655 Villeneuve d’Ascq Cédex France [email protected] Dedicated to Alan Weinstein on the occasion of his 60th birthday. Abstract. Higher homotopy generalizations of Lie–Rinehart algebras, Gerstenhaber, and Batalin–Vilkovisky algebras are explored. These are defined in terms of various antisymmetric bilinear operations satisfying weakened versions of the Jacobi identity, as well as in terms of operations involving more than two variables of the Lie triple systems kind. A basic tool is the Maurer–Cartan algebra—the algebra of alternating forms on a vector space so that Lie brackets correspond to square zero derivations of this algebra—and multialgebra generalizations thereof. The higher homotopies are phrased in terms of these multialgebras. Applications to foliations are discussed: objects which serve as replacements for the Lie algebra of vector fields on the “space of leaves’’ and for the algebra of multivector fields are developed, and the spectral sequence of a foliation is shown to arise as a special case of a more general spectral sequence including the Hodge–de Rham spectral sequence.

Introduction In this paper we will explore, in the framework of Lie–Rinehart algebras and suitable higher homotopy generalizations thereof, various antisymmetric bilinear operations satisfying weakened versions of the Jacobi identity, as well as similar operations involving more than two variables; such operations have recently arisen in algebra, differential geometry, and mathematical physics but are lurking already behind a number of classical developments. Our aim is to somewhat unify these structures by means of the relationship between Lie–Rinehart, Gerstenhaber, and Batalin–Vilkovisky algebras which we first observed in Huebschmann [1998a]. This will be, perhaps, a first step towards taming the bracket zoo that arose recently in topological field theory; see what we wrote in the introduction to Huebschmann [1998a]. The notion of Lie–Rinehart algebra and its generalization are likely to provide a good conceptual

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framework for that purpose. It will also relate new notions like those of Gerstenhaber and Batalin–Vilkovisky algebra, and generalizations thereof, with classical ones like those of connection, curvature, and torsion, as well as with less classical ones like the triple product isolated by Yamaguti [1957–1958] and operations of the kind introduced by Kinyon and Weinstein [2001]; it will connect new developments with old results due to Cartan [1927] and Nomizu [1954] describing the geometry of Lie groups and of reductive homogeneous spaces and, more generally, with more recent results in the geometry of Lie loops; see Kikkawa [1975] and Sabinin and Mikheev [1988]. We will see that the new structures have incarnations of a mathematical nature, e.g., in the theory of foliations. The higher homotopies which are exploited below are of a special kind, where only the first of an (in general) infinite family is nonzero. Let R be a commutative ring with 1. A Lie–Rinehart algebra (A, L) consists of a commutative R-algebra A, an R-Lie algebra L, an A-module structure on L, and an action L ⊗R A → A of L on A by derivations. These are required to satisfy suitable compatibility conditions which arise by abstraction from the pair (A, L) = (C ∞ (M), Vect(M)) consisting of the smooth functions C ∞ (M) and smooth vector fields Vect(M) on a smooth manifold M. A complete definition will be recalled in Section 1 below. In Huebschmann [1990], [1991a], [1998a], [1998b], [1999a], [1999b], [2000], [2001], [2002] we studied these objects and variants thereof and used them to solve various problems in algebra and geometry. See Huebschmann [2003] for a survey and leisurely introduction. In differential geometry, a special case of a Lie–Rinehart algebra arises from the space of sections of a Lie algebroid. In Huebschmann [1998a], [1998b], and [2000] we have shown that certain Gerstenhaber and Batalin–Vilkovisky algebras admit natural interpretations in terms of Lie–Rinehart algebras. The starting point was the following observation: It is nowadays well understood that a skew-symmetric bracket on a vector space g is a Liebracket (i.e., satisfies the Jacobi identity) if and only if the coderivation ∂ on the graded exterior coalgebra [sg] corresponding to the bracket on g has square zero, i.e., is a differential; this coderivation is then the ordinary Lie algebra homology operator. This kind of characterization is not available for a general Lie–Rinehart algebra: Given a commutative algebra A and an A-module L, a Lie–Rinehart structure on (A, L) cannot be characterized in terms of a coderivation on A [sL] with reference to a suitable coalgebra structure on A [sL] (unless the L-action on A is trivial); in fact, in the Lie–Rinehart context, a certain dichotomy between A-modules and chain complexes which are merely defined over R persists thoughout; see, e.g., the Remark 2.5.2 below. On the other hand, Lie–Rinehart algebra structures on (A, L) correspond to Gerstenhaber algebra structures on the exterior A-algebra A [sL]; see, e.g., KosmannSchwarzbach [1995]. In particular, when A is the ground ring and L just an ordinary Lie algebra g, under the obvious identification of [sg] and [sg] as graded Rmodules, the (uniquely determined) generator of the Gerstenhaber bracket on [sg] is exactly the Lie algebra homology operator on [sg]. Given a general commutative algebra A and an A-module L, the interpretation of Lie–Rinehart algebra structures on (A, L) in terms of Gerstenhaber algebra structures on A [sL] provides, among other things, a link between Gerstenhaber [1963] and Rinehart [1963] (which seems

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to have been completely missed in the literature). In the present paper, we will extend this link to suitable higher homotopy notions which we refer to by the attribute “quasi’’; we will introduce Lie–Rinehart triples, quasi-Lie–Rinehart algebras, and certain quasi-Gerstenhaber algebras and quasi-Batalin–Vilkovisky algebras, and we will explore the various relationships between these notions. Below we will comment on the relationship with notions of quasi-Gerstenhaber and quasi-Batalin–Vilkovisky algebras already in the literature. When an algebraic structure (e.g., a commutative algebra, Lie algebra, etc.) is “resolved’’ by an object, which we here somewhat vaguely refer to as a “resolution’’ (free, or projective, or variants thereof) having the given structure as its zero-th homology, on the resolution, the algebraic structure is in general defined only up to higher homotopies; likewise, an A∞ structure is defined in terms of a bar construction or variants thereof; see, e.g., Huebschmann and Kadeishvili [1991], Huebschmann and Stasheff [2002], and the references there. Exploiting higher homotopies of this kind, in a series of articles we constructed small free resolutions for certain classes of groups from which we then were able to do explicit calculations in group cohomology which up to now still cannot be done by other methods; see Huebschmann [1989a], [1989b], [1989c], [1991b]. A historical overview related with A∞ -structures may be found in the Addendum to Keller [2001]; see also Huebschmann [1999c] and Huebschmann and Kadeishvili [1991] for more historical comments. In this paper, we will explore a certain higher homotopy related with Lie–Rinehart algebras and variants thereof. A Lie algebra up to higher homotopies (equivalently: L∞ -algebra) on an R-chain complex h may be defined in terms of a coalgebra perturbation of the differential on the graded symmetric coalgebra on the suspension of h; alternatively, it may be defined in terms of a suitable Maurer–Cartan algebra (see below). Since a genuine Lie–Rinehart structure on (A, L) cannot be characterized in terms of a coderivation on A [sL], the first alternative breaks down for a general Lie–Rinehart algebra. The higher homotopies we will explore in this paper do not live on an object close to a resolution of the above kind or close to a symmetric coalgebra; they may conveniently be phrased in terms of an object of a rather different nature which, extending terminology introduced by van Est [1989], we refer to as a Maurer–Cartan algebra. A special case thereof arises in the following fashion: Given a finite dimensional vector space g over a field k, skew symmetric brackets on g correspond bijectively to degree −1 derivations of the graded algebra of alternating forms on g (with reference to multiplication of forms), and those brackets which satisfy the Jacobi identity correspond to square zero derivations, i.e., differentials. This observation generalizes to Lie–Rinehart algebras of the kind (A, L) under the assumption that L be a finitely generated projective A-module; see Theorem 2.2.16 below. For an ordinary Lie algebra g over a field k, in van Est [1989], the resulting differential graded algebra Alt(g, k) (which calculates the cohomology of g) has been called Maurer– Cartan algebra. The main point of this paper is that higher homotopy variants of the notion of Maurer–Cartan algebra provide the correct framework to phrase certain higher homotopy versions of Lie–Rinehart, Gerstenhaber, and Batalin–Vilkovisky

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algebras to which we will refer to as quasi-Lie–Rinehart-, quasi-Gerstenhaber, and quasi-Batalin–Vilkovisky algebras. The differential graded algebra of alternating forms on a Lie algebra occurs, at least implicitly, in Cartan [1929] and has a long history of use since then (see Koszul [1985]); once I learned in a talk by van Est that this algebra has been used by E. Cartan in the 1930s to characterize the structure of Lie groups and Lie algebras. For the reader’s convenience, we will explain briefly and somewhat informally a special case of a quasi-Lie–Rinehart algebra at the present stage: Let (M, F) be a foliated manifold, the foliation being written as F, let τF be the tangent bundle of the foliation F, and choose a complement ζ of τF so that the tangent bundle τM of M may be written as τM = τF ⊕ ζ . Let LF ⊆ Vect(M) be the Lie algebra of smooth vector fields tangent to the foliation F, and let Q be the C ∞ (M)-module (ζ ) of smooth sections of ζ . The Lie bracket in Vect(M) induces a left LF -module structure on Q—the Bott connection— and the space QLF of invariants, that is, of vector fields on M which are horizontal (with respect to the decomposition τM = τF ⊕ ζ ) and constant on the leaves inherits a Lie bracket. The standard complex A arising from a fine resolution of the sheaf of germs of functions on M which are constant on the leaves acquires a differential graded algebra structure and has H0 (A) equal to the algebra of functions on M which are constant on the leaves, and the Lie algebra QLF of invariants arises as H0 (Q), where Q is the complex coming from a fine resolution of the sheaf VQ of germs of vector fields on M which are horizontal (with respect to the decomposition (τM ) = LF ⊕ Q) and constant on the leaves. In a sense, QLF is the Lie algebra of vector fields on the “space of leaves,’’ that is, the space of sections of a certain geometric object which may be seen as a replacement for the in general nonexistant tangent bundle of the “space of leaves.’’ Within our approach, this philosophy is pushed further in the following fashion: The pair (A, Q) acquires what we will call a quasi-Lie–Rinehart structure in an obvious fashion; see (4.12) and (4.15) below for the details. We view A as the algebra of generalized functions and Q as the generalized Lie algebra of vector fields for the foliation. The pair (H0 (A), H0 (Q)) is necessarily a Lie–Rinehart algebra, and the entire cohomology (H∗ (A), H∗ (Q)) acquires a graded Lie–Rinehart algebra structure. As a side remark, we note that here the resolution of the sheaf VQ is by no means a projective one; indeed, it is a fine resolution of that sheaf, the bracket on Q is not an ordinary Lie(-Rinehart) bracket, in particular, does not satisfy the Jacobi identity, and the entire additional structure is encapsulated in certain homotopies which may conveniently be phrased in terms of a suitable Maurer–Cartan algebra that here arises from the de Rham algebra of M. When the foliation does not come from a fiber bundle, the structure of the graded Lie–Rinehart algebra (H∗ (A), H∗ (Q)) will in general be more complicated than in the case when the foliation comes from a fiber bundle. Thus the cohomology of a quasi-Lie–Rinehart algebra involves an ordinary Lie–Rinehart algebra in degree zero but in general contains considerably more information. In particular, in the case of a foliation it contains more than just “functions and vector fields on the space of leaves’’; the additional information partly includes the history of


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the “space of leaves,’’ that is, it includes information as to how this space arises from the foliation, how the leaves sit inside the ambient space, about singularities, etc. In Section 6 we will show that, when the foliation is transversely orientable with a basic transverse volume form ω, a corresponding quasi-Batalin–Vilkovisky algebra isolated in Theorem 6.10 below has an underlying quasi-Gerstenhaber algebra which, in turn, yields a kind of generalized Schouten algebra (generalized algebra of multivector fields) for the foliation; the cohomology of this quasi-Gerstenhaber algebra may then be viewed as the Schouten algebra for the “space of leaves.’’ See (6.15) below for details. Thus our approach will provide new insight, for example, into the geometry of foliations; see in particular (1.12), (2.10), (4.15), (6.15) below. The formal structure behind foliations which we will phrase in terms of quasi-Lie–Rinehart algebras and its offspring does not seem to have been noticed in the literature before—indeed, it involves, among a number of other things, a suitable grading which seems unfamiliar in the literature on quasi-Gerstenhaber and quasi-Batalin–Vilkovisky algebras (see (6.17) below)—or the formal connections with Yamaguti’s triple product and with Lie loops. A simplified version of the question we will examine is this: Given a Lie algebra g with a decomposition g = h ⊕ q, where h is a Lie subalgebra, what kind of structure does q then inherit? Variants of this question and possible answers may be found in a number of places in the literature; see, e.g., Cartan [1927], Nomizu [1954], where, in particular, in a global situation, an answer is given for reductive homogeneous spaces. In the framework of Lie–Rinehart algebras, this issue does not seem to have been raised yet, not even for the special case of Lie algebroids. As a by-product, we find a certain formal relationship between Yamaguti’s triple product and certain forms ∗∗ which may be found in Koszul [1985]. In particular, the failure of a quasi-Gerstenhaber bracket to satisfy the Jacobi identity is measured by an additional piece of structure which we refer to as an h-Jacobiator; an h-Jacobiator, in turn, is defined in terms of Koszul’s forms 3∗ . Likewise, the quadruple and quintuple products studied in Section 3 below are related with Koszul’s forms, and these, in turn, are related with certain higher order operations which may be found, e.g., in Sabinin and Mikheev [1988]. We do not pursue this here; we hope to eventually come back to it in another article. A Courant algebroid has been shown in Roytenberg and Weinstein [1998] to acquire an L∞ -structure, that is, a Lie algebra structure up to higher homotopies. The present paper paves, perhaps, the way towards finding a higher homotopy Lie– Rinehart or higher homotopy Lie algebroid structure on a Courant algebroid incorporating the Courant algebroid structure. Graded quasi-Batalin–Vilkovisky algebras have already been explored in Getzler [1995]. Our notions of quasi-Gerstenhaber and quasi-Batalin–Vilkovisky algebra, while closely related, do not coincide with those in Bangoura [2003], Bangoura [2002], Getzler [1995], Kosmann-Schwarzbach [2005], Roytenberg [2002]. In particular, our algebras are bigraded while those in the cited references are ordinary graded algebras; the appropriate totalization (forced, as noted above, by our application of the newly developed algebraic structure to foliations and written in Section 6 below

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as the functor Tot) of our bigraded objects leads to differential graded objects which are not equivalent to those in the quoted references. See Remark 6.17 below for more details on the relationship between the various notions. Also the approaches differ in motivation; the guiding idea behind Getzler [1995] and Kosmann-Schwarzbach [2005] seems to be Drinfeld’s quasi-Hopf algebras. Our motivation, as indicated above, comes from foliations and the search for appropriate algebraic notions encapsulating the infinitesimal structure of the “space of leaves’’ and its history, as well as the search for a corresponding Lie–Rinehart generalization of the operations on a reductive homogenous space isolated by Nomizu and elaborated upon by Yamaguti (mentioned earlier) and taken up again by Kinyon and Weinstein [2001]. Indeed, this paper was prompted by the preprint versions of Kinyon and Weinstein [2001] and Weinstein [2000]. It is a pleasure to dedicate it to Alan Weinstein.

1 Lie–Rinehart triples Let R be a commutative ring with 1, not necessarily a field; R could be, for example, the algebra of smooth functions on a smooth manifold; see Huebschmann [1999b]. Furthermore, let A be a commutative R-algebra. An (R, A)-Lie algebra (see Rinehart [1963]) is a Lie algebra L over R which acts on (the left of) A (by derivations) and is also an A-module satisfying the compatibility conditions [α, aβ] = α(a)β + a[α, β], (aα)(b) = a(α(b)), where a, b ∈ A and α, β ∈ L and where the operations of A on L and of L on A are written in terms of elements in the obvious fashion. When the emphasis is on the pair (A, L) with the mutual structure of interaction between A and L, we refer to the pair (A, L) as a Lie–Rinehart algebra. Given an ordinary Lie algebra g over R, the pair (R, g) is a Lie–Rinehart algebra in an obvious fashion. Given a smooth foliated manifold, when A denotes the algebra of smooth functions and H the Lie algebra of vector fields tangent to the foliation, the pair (A, H ) is a Lie–Rinehart algebra; under such circumstances it may be convenient to take a ground ring R larger than the reals; for example when the foliation comes from a fiber bundle, for certain problems (e.g., related with duality), the appropriate ground ring is the algebra of smooth functions on the base manifold; see Huebschmann [1999b]. More details and additional references may be found in our survey paper Huebschmann [2003]. The problem we wish to explore is the following. Question 1.1. Given a Lie–Rinehart algebra (A, L) and an A-module direct sum decomposition L = H ⊕ Q inducing an (R, A)-Lie algebra structure on H , what kind of structure does Q then inherit, and by what additional structure are H and Q related? Question 1.2. Given an (R, A)-Lie algebra structure on H and the (new) structure (which we will isolate below) on Q, what kind of additional structure turns the A-


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module direct sum L = H ⊕ Q into an (R, A)-Lie algebra in such a way that the latter induces the given structure on H and Q? Example 1.3.1. Let g be an ordinary R-Lie algebra with a decomposition g = h ⊕ q, where h is a Lie subalgebra. Recall that the decomposition of g is said to be reductive (see Nomizu [1954]) provided [h, q] ⊆ q. Such a reductive decomposition arises from a reductive homogeneous space; see Cartan [1927], Kikkawa [1975], Nomizu [1954], Sabinin and Mikheev [1988], Yamaguti [1957–1958]. For example, every homogeneous space of a compact Lie group or, more generally, of a reductive Lie group, is reductive. Nomizu [1954] has shown that on such a reductive homogeneous space, the torsion and curvature of the “canonical affine connection of the second kind’’ (affine connection with parallel torsion and curvature) yield a bilinear and a ternary operation which, at the identity, come down to a certain bilinear and ternary operation on the constituent q; Yamaguti [1957–1958] gave an algebraic characterization of pairs of such operations. Example 1.3.2. A quasi-Lie bialgebra (h, q) (see Kosmann-Schwarzbach [1992]) consists of a (real or complex) Lie algebra h and a (real or complex) vector space q with suitable additional structure where q = h∗ , so that g = h ⊕ h∗ is an ordinary Lie algebra; the pair (g, h) is occasionally referred to in the literature as a Manin pair. Quasi-Lie bialgebras arise as classical limits of quasi-Hopf algebras; these, in turn, were introduced by Drinfeld [1990]. Example 1.4.1. Let R be the field R of real numbers, let (M, F) be a foliated manifold, let τF be the tangent bundle of the foliation F, and choose a complement ζ of τF so that the tangent bundle τM of M may be written as τM = τF ⊕ ζ . Thus, as a vector bundle, ζ is canonically isomorphic to the normal bundle of the foliation. Let (A, L) be the Lie–Rinehart algebra (C ∞ (M), Vect(M)), let H = LF ⊆ L be the (R, A)-Lie algebra of smooth vector fields tangent to the foliation F, and let Q be the A-module (ζ ) of smooth sections of ζ . Then L = H ⊕ Q is an A-module direct sum decomposition of the (R, A)-Lie algebra L, and the question arises as to what kind of Lie structure Q carries. This question, in turn, may be subsumed under the more general question to what extent the “space of leaves’’ can be viewed as a smooth manifold. This more general question is not only of academic interest since, for example, in certain physical situations, the true classical state space of a constrained system is the “space of leaves’’ of a foliation which is in general not fibrating, and the Noether theorems are conveniently phrased in the framework of foliations. Example 1.4.2. Let R be the field C of complex numbers, M a smooth complex manifold M, A the algebra of smooth complex functions on M, L the (C, A)-Lie algebra of smooth complexified vector fields, and let L and L be the spaces of smooth sections of the holomorphic and antiholomorphic tangent bundle of M, respectively. Then L and L are (C, A)-Lie algebras, and (A, L , L ) is a twilled Lie–Rinehart algebra in the sense of Huebschmann [1998b], Huebschmann [2000]. Adjusting the notation to that in Example 1.4.1, let H = L and Q = L . Thus, in this particular case, Q = L is in fact an ordinary (R, A)-Lie algebra, and the additional structure

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relating H and Q is encapsulated in the notion of twilled Lie–Rinehart algebra. The integrability condition for an almost complex structure may be phrased in terms of the twilled Lie–Rinehart axioms; see Huebschmann [1998b], Huebschmann [2000] for details. The situation of Example 1.4.1 is somewhat more general than that of Example 1.4.2 since in Example 1.4.1 the constituent Q carries a structure which is more general than that of an ordinary (R, A)-Lie algebra. Another example for a decomposition of the kind spelled out in Questions 1.1 and 1.2 above arises from combining the situations of Example 1.4.1 and of Example 1.4.2, that is, from a smooth manifold foliated by holomorphic manifolds, and yet another example arises from a holomorphic foliation. Abstracting from these examples, we isolate the notion of a Lie–Rinehart triple. For ease of exposition, we also introduce the weaker concepts of almost preLie–Rinehart triple and pre-Lie–Rinehart triple. Distinguishing among these three notions may appear pedantic but will clarify the statement of Theorem 2.7 below. See also Remark 2.8.4 below. Our usage of the term triple (to be isolated below) is not consistent with that of Manin triple in the literature. A Lie–Rinehart algebra involves a pair consisting of an algebra and a Lie algebra; in this context, it is also common in the literature to refer to this kind of structure as a pair (see Huebschmann [2003] for more details), and this usage of the term pair, in turn, is not consistent with the notion of a Manin pair. Below we will consider triples involving a commutative algebra A and two A-modules H and Q, just as in Example 1.4.1 and Example 1.4.2 above, and (A, H ⊕ Q) will be a Lie–Rinehart algebra if and only if (A, H, Q) is a Lie–Rinehart triple (so far unexplained). These remarks are intended to justify our terminology Lie–Rinehart triple. We now proceed towards the description of Lie–Rinehart triples. Let A be a commutative R-algebra. Consider two A-modules H and Q, together with • • •

skew-symmetric R-bilinear brackets of the kind (1.5.1.H ) and (1.5.1.Q) below, not necessarily Lie brackets; R-bilinear operations of the kind (1.5.2.H ), (1.5.2.Q), (1.5.3), (1.5.4) below; and a skew-symmetric A-bilinear pairing δ of the kind (1.5.5) below: [·, ·]H : H ⊗R H − → H, → Q, [·, ·]Q : Q ⊗R Q − H ⊗R A − → A, x ⊗R a → x(a), Q ⊗R A − → A, ξ ⊗R a → ξ(a), → Q, · : H ⊗R Q − · : Q ⊗R H − → H, δ : Q ⊗A Q − → H.

(1.5.1.H ) (1.5.1.Q) x ∈ H, a ∈ A,

(1.5.2.H )

ξ ∈ Q, a ∈ A,

(1.5.2.Q) (1.5.3) (1.5.4) (1.5.5)

We will say that the data (A, H, Q) constitute an almost pre-Lie–Rinehart triple provided they satisfy (i), (ii), and (iii) below.


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(i) The values of the adjoints H → End R (A) and Q → End R (A) of (1.5.2.H ) and (1.5.2.Q) respectively lie in Der R (A); (ii) (1.5.1.H ), (1.5.2.H ) and the A-module structure on H and, likewise, (1.5.1.Q), (1.5.2.Q) and the A-module structure on Q, satisfy the following Lie–Rinehart axioms (1.5.6.H ), (1.5.7.H ), (1.5.6.Q), (1.5.7.Q): (ax)(b) = a(x(b)), a, b ∈ A, x ∈ H, [x, ay]H = x(a)y + a[x, y]H , a ∈ A, x, y ∈ H, (aξ )(b) = a(ξ(b)), a, b ∈ A, ξ ∈ Q, [ξ, aη]Q = ξ(a)η + a[ξ, η]Q , a ∈ A, ξ, η ∈ Q;

(1.5.6.H ) (1.5.7.H ) (1.5.6.Q) (1.5.7.Q)

(iii) (1.5.3) and (1.5.4) behave like connections, that is, for a ∈ A, x ∈ H, ξ ∈ Q, the identities x · (aξ ) = (x(a))ξ + a(x · ξ ), (ax) · ξ = a(x · ξ ),

(1.5.8) (1.5.9)

ξ · (ax) = (ξ(a))x + a(ξ · x), (aξ ) · x = a(ξ · x),

(1.5.10) (1.5.11)

are required to hold. We will say that an almost pre-Lie–Rinehart triple (A, H, Q) is a pre-Lie–Rinehart triple provided that (i) (A, H ), endowed with the operations (1.5.1.H ) and (1.5.2.H ), is a Lie–Rinehart algebra—equivalently, the bracket (1.5.1.H ) satisfies the Jacobi identity—, and that (ii) the operation (1.5.3) turns Q into a left (A, H )-module, that is, the “connection’’ given by this operation is “flat,’’ i.e., satisfies the identity [x, y]H · ξ = x · (y · ξ ) − y · (x · ξ ),

x, y ∈ H, ξ ∈ Q.

(1.5.12)

(1.5.13) Thus a pre-Lie–Rinehart triple (A, H, Q) consists of a Lie–Rinehart algebra (A, H ) (the structure of which is given by (1.5.1.H ), (1.5.2.H )) and a left (A, H )module Q (given by the operation (1.5.3) which, in turn, is required to satisfy the axioms (1.5.8) and (1.5.9)) together with the additional structure (1.5.1.Q), (1.5.2.Q), (1.5.4), (1.5.5) subject to the axioms (1.5.6.Q), (1.5.7.Q), (1.5.10), (1.5.11). Given an almost pre-Lie–Rinehart triple (A, H, Q), let L = H ⊕ Q be the Amodule direct sum, and define an R-bilinear skew-symmetric bracket →L [·, ·] : L ⊗R L −

(1.6.1)

by means of the formula [(x, ξ ), (y, η)] = [x, y]H + [ξ, η]Q + δ(ξ, η) + x · η − η · x + ξ · y − y · ξ (1.6.2) and, furthermore, an operation →A L ⊗R A −

(1.6.3)

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in the obvious way, that is, by means of the association (ξ, x) ⊗R a → ξ(a) + x(a),

x ∈ H, ξ ∈ Q, a ∈ A.

(1.6.4)

By construction, the values of the adjoint of (1.6.3) then lie in Der R (A), that is, this adjoint is then of the form L=H ⊕Q− → Der R (A).

(1.6.5)

An almost pre-Lie–Rinehart triple (A, H, Q) will be said to be a Lie–Rinehart triple if (1.6.1) and (1.6.3) turn (A, L), where L = H ⊕ Q, into a Lie–Rinehart algebra. A Lie–Rinehart triple (A, H, Q), where δ is zero, is a twilled Lie–Rinehart algebra in the sense of Huebschmann [1998b], Huebschmann [2000]. Thus Lie–Rinehart triples generalize twilled Lie–Rinehart algebras. A direct sum decomposition L = H ⊕ Q of an (R, A)-Lie algebra L such that (A, H ) inherits a Lie–Rinehart structure yields a Lie–Rinehart triple (A, H, Q) in an obvious fashion: The brackets (1.5.1.H ) and (1.5.1.Q) result from restriction and projection; the operations (1.5.2.H ) and (1.5.2.Q) are obtained by restriction as well; further, the requisite operations (1.5.3) and (1.5.4) are given by the composites [·,·]|H ⊗R Q

prQ

[·,·]|Q⊗R H

prH

· : H ⊗R Q −−−−−−→ H ⊕ Q −−→ Q and

· : Q ⊗R H −−−−−−→ H ⊕ Q −−→ H,

(1.7.1)

(1.7.2)

where, for M = H ⊗R Q and M = Q ⊗R H , [·, ·]|M denotes the restriction of the Lie bracket to M. The pairing (1.5.5) is the composite [·,·]|Q⊗R Q

prH

δ : Q ⊗A Q −−−−−−→ L = H ⊕ Q −−→ H ;

(1.7.3)

at first it is only R-bilinear but is readily seen to be A-bilinear. The formula (1.6.2) is then merely a decomposition of the initially given bracket on L into components according to the direct sum decomposition of L into H and Q, and (1.6.3) is accordingly a decomposition of the L-action on A. Furthermore, given x, y ∈ H and ξ ∈ Q, in L we have the identity [x, y] · ξ − ξ · [x, y] = [[x, y], ξ ] = [x, [y, ξ ]] − [y, [x, ξ ]] = x · (y · ξ ) − (y · ξ ) · x − [x, ξ · y] − y · (x · ξ ) + (x · ξ ) · y − [ξ · x, y] which at once implies (1.5.12). Remark 1.8.1. Thus we see that, in particular, if an almost pre-Lie–Rinehart triple (A, H, Q) is a Lie–Rinehart triple, it is necessarily a pre-Lie–Rinehart triple; see (1.5.13). Remark 1.8.2. In the situation of Example 1.3.2, when g arises from a quasi-Lie bialgebra (so that q = h∗ ), in the literature, the piece of structure δ is often written as an element of 3 h.


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Theorem 1.9. A pre-Lie–Rinehart triple (A, H, Q) is a genuine Lie–Rinehart triple, that is, the bracket [·, ·] (see (1.6.1)) and the operation (1.6.3) turn (A, L), where L = H ⊕ Q, into a Lie–Rinehart algebra, if and only if the brackets [·, ·]H and [·, ·]Q on H and Q, respectively, and the operations (1.5.3), (1.5.4), and (1.5.5), are related by ξ(x(a)) − x(ξ(a)) = (ξ · x)(a) − (x · ξ )(a), x · [ξ, η]Q = [x · ξ, η]Q + [ξ, x · η]Q − (ξ · x) · η + (η · x) · ξ, ξ · [x, y]H = [ξ · x, y]H + [x, ξ · y]H

(1.9.1) (1.9.2)

− (x · ξ ) · y + (y · ξ ) · x,

(1.9.3)

ξ(η(a)) − η(ξ(a)) = [ξ, η]Q (a) + (δ(ξ, η))(a),

(1.9.4)

[ξ, η]Q · x = ξ · (η · x) − η · (ξ · x) − δ(x · ξ, η) − δ(ξ, x · η) + [x, δ(ξ, η)]H , [[ξ, η]Q , ϑ]Q + (δ(ξ, η)) · ϑ = 0,

(ξ,η,ϑ) cyclic

δ([ξ, η]Q , ϑ) =

(ξ,η,ϑ) cyclic

ξ · δ(η, ϑ),

(1.9.5) (1.9.6) (1.9.7)

(ξ,η,ϑ) cyclic

where a ∈ A, x, y ∈ H , ξ, η, ϑ ∈ Q. Recall that given a commutative algebra A and Lie–Rinehart algebras (A, L ), (A, L) and (A, L ), where L is an ordinary A-Lie algebra, an extension of Lie– Rinehart algebras 0− → L − →L− → L − →0 is an extension of A-modules which is also an extension of ordinary Lie algebras so that the projection from L to L is a morphism of Lie–Rinehart algebras; see Huebschmann [1999a]. Theorem 1.9 entails at once the following. Corollary 1.9.8. Given a Lie–Rinehart triple (A, H, Q), the left (A, H )-module structures (1.5.2.H ) on A and (1.5.3) on Q are trivial if and only if (A, Q) is a Lie– Rinehart algebra in such a way that the projection from E = H ⊕ Q to Q fits into an extension 0− →H − →E− →Q− →0 of Lie–Rinehart algebras. Thus Lie–Rinehart triples (A, H, Q) having trivial left (A, H )-module structures on A and Q and extensions of Lie–Rinehart algebras of the kind (A, L) together with an A-module section of the projection map are equivalent notions. Proof of Theorem 1.9. The bracket (1.6.1) is plainly skew-symmetric. Hence the proof comes down to relating the Jacobi identity in L and the Lie–Rinehart compatibility properties with (1.9.1)–(1.9.7).

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Thus, suppose that the bracket [·, ·] on L = H ⊕ Q given by (1.6.1) and the operation L ⊗R A → A given by (1.6.3) turn (A, L) into a Lie–Rinehart algebra. Given ξ ∈ Q and x ∈ H , we have [ξ, x] = ξ · x − x · ξ ; since L acts on A by derivations, for a ∈ A, we conclude that ξ(x(a)) − x(ξ(a)) = [ξ, x](a) = (ξ · x)(a) − (x · ξ )(a), that is, (1.9.1) holds. Likewise, given ξ, η ∈ Q, [ξ, η] = [ξ, η]Q + δ(ξ, η) ∈ L, whence, for a ∈ A, ξ(η(a)) − η(ξ(a)) = [ξ, η](a) = [ξ, η]Q (a) + (δ(ξ, η))(a), that is, (1.9.4) holds. Next, since L is a Lie algebra, its bracket satisfies the Jacobi identity. Hence, given x ∈ H and ξ, η ∈ Q, x · [ξ, η]Q − [ξ, η]Q · x = [x, [ξ, η]Q ] = [x, [ξ, η]] − [x, δ(ξ, η)] = [[x, ξ ], η] + [ξ, [x, η]] − [x, δ(ξ, η)] = [x · ξ − ξ · x, η] + [ξ, x · η − η · x] − [x, δ(ξ, η)]H = [x · ξ, η] − [ξ · x, η] + [ξ, x · η] − [ξ, η · x] − [x, δ(ξ, η)]H = [x · ξ, η] + [ξ, x · η] − (ξ · x) · η + η · (ξ · x) + (η · x) · ξ − ξ · (η · x) − [x, δ(ξ, η)]H = [x · ξ, η]Q + δ(x · ξ, η) + [ξ, x · η]Q + δ(ξ, x · η) − (ξ · x) · η + η · (ξ · x) + (η · x) · ξ − ξ · (η · x) − [x, δ(ξ, η)]H , whence, comparing components in H and Q, we conclude that x · [ξ, η]Q = [x · ξ, η]Q + [ξ, x · η]Q − (ξ · x) · η + (η · x) · ξ, [ξ, η]Q · x = ξ · (η · x) − η · (ξ · x) − δ(x · ξ, η) − δ(ξ, x · η) + [x, δ(ξ, η)]H , that is, (1.9.2) and (1.9.5) hold. Likewise, given ξ ∈ Q and x, y ∈ H , ξ · [x, y]H − [x, y]H · ξ = [ξ, [x, y]H ] = [[ξ, x], y] + [x, [ξ, y]] = [ξ · x − x · ξ, y] + [x, ξ · y − y · ξ ] = [ξ · x, y] − [x · ξ, y] + [x, ξ · y] − [x, y · ξ ] = [ξ · x, y] + [x, ξ · y] − (x · ξ ) · y + y · (x · ξ ) + (y · ξ ) · x − x · (y · ξ ) = [ξ · x, y]H + [x, ξ · y]H − (x · ξ ) · y + y · (x · ξ ) + (y · ξ ) · x − x · (y · ξ ),


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whence, comparing components in Q and H , we conclude that ξ · [x, y]H = [ξ · x, y]H + [x, ξ · y]H − (x · ξ ) · y + (y · ξ ) · x [x, y]H · ξ = x · (y · ξ ) − y · (x · ξ ), that is, (1.9.3) and (1.5.12) hold; notice that (1.5.12) holds already by assumption. Next, given ξ, η, ϑ ∈ Q, [[ξ, η], ϑ] = [[ξ, η]H , ϑ] + [[ξ, η]Q , ϑ] = [δ(ξ, η), ϑ] + [[ξ, η]Q , ϑ] = [δ(ξ, η), ϑ]H + [δ(ξ, η), ϑ]Q + [[ξ, η]Q , ϑ]H + [[ξ, η]Q , ϑ]Q = (δ(ξ, η)) · ϑ − ϑ · δ(ξ, η) + δ([ξ, η]Q , ϑ) + [[ξ, η]Q , ϑ]Q . Hence [[ξ, η], ϑ] + [[η, ϑ], ξ ] + [[ϑ, ξ ], η] = (δ(ξ, η)) · ϑ + (δ(η, ϑ)) · ξ + (δ(ϑ, ξ )) · η + [[ξ, η]Q , ϑ]Q + [[η, ϑ]Q , ξ ]Q + [[ϑ, ξ ]Q , η]Q − ξ · δ(η, ϑ) − η · δ(ϑ, ξ ) − ϑ · δ(ξ, η) + δ([ξ, η]Q , ϑ) + δ([η, ϑ]Q , ξ ) + δ([ϑ, ξ ]Q , η). Thus the Jacobi identity implies that [[ξ, η]Q , ϑ]Q + [[η, ϑ]Q , ξ ]Q + [[ϑ, ξ ]Q , η]Q +(δ(ξ, η)) · ϑ + (δ(η, ϑ)) · ξ + (δ(ϑ, ξ )) · η = 0 δ([ξ, η]Q , ϑ) + δ([η, ϑ]Q , ξ ) + δ([ϑ, ξ ]Q , η) −ξ · δ(η, ϑ) − η · δ(ϑ, ξ ) − ϑ · δ(ξ, η) = 0, that is, (1.9.6) and (1.9.7) are satisfied. Conversely, suppose that the brackets [·, ·]H and [·, ·]Q on H and Q, respectively, and the operations (1.5.3), (1.5.4), and (1.5.5), are related by (1.9.1)–(1.9.7). We can then read the above calculations backwards and conclude that the bracket (1.6.1) on L satisfies the Jacobi identity and the operation (1.6.3) yields a Lie algebra action of L on A by derivations. The remaining Lie–Rinehart algebra axioms hold by assumption. Thus (A, L) is a Lie–Rinehart algebra.

Remark 1.10. Under the circumstances of Example 1.3, the requirements (1.5.6.Q), (1.5.6.H ), (1.5.7.Q), (1.5.7.H ), (1.5.8)–(1.5.11) are vacuous, and so are (1.9.1) and (1.9.4) as well. Given an (R, A) Lie algebra L and an (R, A) Lie subalgebra H , the invariants AH ⊆ A constitute a subalgebra of A; we will then denote the normalizer of H in L in the sense of Lie algebras by LH , that is, LH consists of all α ∈ L having the property that [α, β] ∈ H whenever β ∈ H .

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Corollary 1.11. Given a Lie–Rinehart triple (A, H, Q), the corresponding (R, A)Lie algebra being written as L = H ⊕ Q, the intersection Q ∩ LH coincides with the invariants QH under the H -action on Q (given by the corresponding operation (1.5.3)), the pair (AH , QH ) acquires a Lie–Rinehart algebra structure, and the projection from LH to QH fits into an extension 0− →H − → LH − → QH − →0

(1.11.1)

of (R, AH )-Lie algebras. Furthermore, the restriction of δ to QH is a cocycle for this extension, that is, it yields the curvature of the connection for the extension determined by the AH -module direct sum decomposition LH = H ⊕ QH . Notice that H is here viewed as an ordinary AH -Lie algebra, the H -action on AH being trivial by construction. Proof . Indeed, given α ∈ Q and β ∈ H , [α, β] = α · β − β · α ∈ L, whence [α, β] ∈ H for every β ∈ H if and only if β · α = 0 ∈ Q for every β ∈ H , that is, if and only if α is invariant under the H -action on Q. The rest of the claim is an immediate consequence of Theorem 1.9.

Illustration 1.12. Under the circumstances of Example 1.4.1, Corollary 1.11 obtains, with H = LF . Now AH = ALF ⊆ A is the algebra of smooth functions which are constant on the leaves, that is, the algebra of functions on the “space of leaves,’’ and LH consists of the vector fields which “project’’ to the “space of leaves.’’ Indeed, given a function f which is constant on the leaves and vector fields X ∈ LH and Y ∈ LF , necessarily Y (Xf ) = [Y, X]f + X(Yf ) = 0, whence Xf is constant on the leaves as well. Thus we may view QH as the Lie algebra of vector fields on the “space of leaves,’’ that is, as the space of sections of a certain geometric object which serves as a replacement for the in general nonexistant tangent bundle of the “space of leaves.’’ Remark 1.13. In analogy with the deformation theory of complex manifolds, given a Lie–Rinehart triple (A, H, Q), we may view H and Q as corresponding to the antiholomorphic and holomorphic tangent bundle, respectively, and accordingly study deformations of the Lie–Rinehart triple via morphisms ϑ : H → Q and spell out the resulting infinitesimal obstructions. This will include a theory of deformations of foliations. Details will be given elsewhere.

2 Lie–Rinehart triples and Maurer–Cartan algebras In this section we will explore the relationship between Lie–Rinehart triples and suitably defined Maurer–Cartan algebras. In particular, we will show that, under an additional assumption, the two notions are equivalent; see Theorem 2.8.3 below for details. As an application we will explain how the spectral sequence of a foliation and the Hodge–de Rham spectral sequence arise as special cases of a single conceptually simple construction. More applications will be given in subsequent sections.


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2.1. Maurer–Cartan algebras Given an A-module L and an R-derivation d of degree −1 on the graded A-algebra Alt A (L, A), we will refer to (Alt A (L, A), d) as a Maurer–Cartan algebra (over L) provided d has square zero, i.e., is a differential. Recall that a multicomplex (over R) is a bigraded R-module {M p,q }p,q together with an operator dj : M p,q → M p+j,q−j +1 for every j ≥ 0 such that the sum d = d0 + d1 + . . . is a differential, i.e., dd = 0; under such circumstances, an infinite sequence of operators of the kind (d2 , d3 , . . . ) is a system of higher homotopies. We will refer to a multicomplex (M; d0 , d1 , d2 , . . . ) whose underlying bigraded object M is endowed with a bigraded algebra structure such that the operators dj are derivations with respect to this algebra structure as a multialgebra and, when it is necessary to spell out the ground ring explicitly, we will refer to a multi-R-algebra. The idea of multicomplex already occurs in Heller [1954], Liulevicius [1963], Wall [1961] and was exploited in various other places in the literature including Huebschmann [1989c], Huebschmann [1991b]. The terminology multicomplex goes back at least to unpublished mimeographed notes of Liulevicius from the 1960s. Given A-modules H and Q, consider the bigraded A-algebra (Alt A (Q, Alt A (H, A)); we will refer to a multi-R-algebra structure (beware: not multi-A-algebra structure) on this bigraded A-algebra having at most d0 , d1 , d2 nonzero as a Maurer–Cartan algebra structure. The resulting multi-R-algebra will then be written as (Alt A (Q, Alt A (H, A)); d0 , d1 , d2 )

(2.1.1)

and referred to as a (multi-)Maurer–Cartan algebra (over (Q, H )). Usually we will discard “multi’’ and more simply refer to a Maurer–Cartan algebra. We note that, for degree reasons, when (2.1.1) is a Maurer–Cartan algebra, the operator d2 is necessarily an A-derivation (since d2 (a) = 0 for every a ∈ A ∼ = Alt 0A (Q, Alt 0A (H, A))). Remark 2.1.2. In this definition, we could allow for nonzero derivations of the kind dj for j ≥ 3 as well. This would lead to a more general notion of multi-Maurer– Cartan algebra not studied here. The presence of a nonzero operator at most of the kind d2 is an instance of a higher homotopy of a special kind which suffices to explain the “quasi’’ structures explored later in the paper. Remark 2.1.3. Given a (multi-)Maurer–Cartan algebra of the kind (2.1.1), the sum d = d0 + d1 + d2 turns Alt A (Q ⊕ H, A) into a Maurer–Cartan algebra. However, not every Maurer–Cartan structure on Alt A (Q ⊕ H, A) arises in this fashion, that is, a multi-Maurer–Cartan algebra structure captures additional structure of interaction between A, Q, and H , indeed, it captures essentially a Lie–Rinehart triple structure. The purpose of the present section is to make this precise. For later reference, we spell out the following, the proof of which is immediate.

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Proposition 2.1.4. Given the three derivations d0 , d1 , d2 , (Alt ∗A (Q, Alt ∗A (H, A)), d0 , d1 , d2 ) is a (multi-)Maurer–Cartan algebra if and only if the following identities are satisfied. d0 d0 = 0

(2.1.4.1)

d0 d1 + d1 d0 = 0 d0 d2 + d1 d1 + d2 d0 = 0 d1 d2 + d2 d1 = 0

(2.1.4.2)

d2 d2 = 0.

(2.1.4.5)

(2.1.4.3) (2.1.4.4)

2.2. Lie–Rinehart and Maurer–Cartan algebras Let A be a commutative R-algebra and L an A-module, together with a skewsymmetric R-bilinear bracket [·, ·]L : L ⊗R L − →L

(2.2.1)

and an operation L ⊗R A − → A,

x ⊗R a → x(a),

x ∈ H, a ∈ A

(2.2.2)

such that the values of the adjoint L − → End R (A) lie in Der R (A) and that (2.2.1), (2.2.2) and the A-module structure on L satisfy the Lie–Rinehart axioms (2.2.3) and (2.2.4) below: (ax)(b) = a(x(b)), a, b ∈ A, x ∈ L, [x, ay]L = x(a)y + a[x, y]L , a ∈ A, x, y ∈ L.

(2.2.3) (2.2.4)

Let M be a graded A-module, together with an operation L ⊗R M − → M,

x ⊗ m → x(m),

x ∈ L, m ∈ m

(2.2.5)

subject to the following requirement: For α ∈ L, a ∈ A, m ∈ M, (aα)(m) = a(α(m)), α(am) = aα(m) + α(a)m.

(2.2.6) (2.2.7)

We refer to an operation of the kind (2.2.5) as a generalized L-connection on M. Under these circumstances, the ordinary Cartan–Chevalley–Eilenberg (CCE) operator d is defined, at first on the bigraded object AltR (L, M) of M-valued R-multilinear alternating forms on L. Indeed, given an R-multilinear alternating function f on L of n − 1 variables which is homogeneous, i.e., the values of f lie in a homogeneous constituent of M, the Cartan–Chevalley–Eilenberg (CCE) formula yields

Homotopies and Maurer–Cartan algebras n

(−1)|f |+1 (df )(α1 , . . . , αn ) = +

253

(−1)(i−1) αi (f (α1 , . . . α=i . . . , αn ))

i=1

(−1)(j +k) f ([αj , αk ], α1 , . . . α=j . . . α=k . . . , αn ),

1≤j 0}. It will be convenient to denote the subtorus of T perpendicular to I by T I . Assume that (M, ω) carries a Hamiltonian T action with moment map µ. For simplicity assume that the T action is effective so that µ(M) is a polytope of dimension equal to dim T . As a topological space the symplectic cut with respect to a cone = β is the space M = µ−1 ()/ ∼, where x ∼ x if µ(x) = µ(x ) ∈ βI and x and x lie in the same T I orbit. Clearly, the torus action on M descends to an action on M . Notice that the action on M is not effective unless dim = dim T , since the subtorus T of T perpendicular to acts trivially on M . In the case of a circle action, when every cone is just a ray, Lerman [Le] realized that under certain mild conditions this space is an orbifold, it carries a natural symplectic form, and the residual torus action is Hamiltonian. As shown in [LMTW] similar results hold for symplectic cuts with respect to cones. Even more generally, symplectic cutting has been extended to cutting with respect to polytopes [LMTW], cutting for nonabelian groups [Me] and Kähler cutting with respect to polytopes [BGL]. For the purposes of this paper we only need to consider symplectic cutting with respect to cones. To recall the results of [LMTW] let us give another construction of M . Let Cβi be a complex line on which T acts with weight βi . Let Cβ = Cβ1 × · · · × Cβk . Then the T action on Cβ is Hamiltonian with respect to the symplectic form ωC = √ −1 dzi ∧ d z¯ i , where zi is the standard complex coordinate on Cβi . Its moment map is ψ(z) = βi |zi |2 , so that the image of Cβ under the moment map is the cone . Consider the symplectic form (ω, −ωC ) on M × Cβ . Then the diagonal torus T ⊂ T × T acts on this space in a Hamiltonian fashion and its moment map φ is given by φ(x, z) = µ(x) − ψ(z). As shown in [LMTW] the symplectic cut M is homeomorphic to the symplectic reduction (M × Cβ )//0 T . Hence, to guarantee that M is a symplectic orbifold it is enough to assume that zero is a regular value of φ. It is easy to see that this is equivalent to the following:

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(*) Every I is transverse to every wall W of µ(M), that is, dim( I ∩ W ) ≤ |I | + dim W − dim T . If (*) holds, we say that is transverse to µ and from now on we consider only the cones satisfying (*). We can write T × T as the product of the first copy of T (that is, T × e) and T . Hence after reducing M × Cβ with respect to T , the action of the first copy of T descends to an action on the reduction M . As shown in [LMTW], this action is Hamiltonian and there exists a moment map µ on M whose image is the intersection µ(M) ∩ . Let us describe the connected components of the fixed point set MT . We will separate them into three sets: the old fixed points, the new fixed points, and the fixed points at zero. Definition 2.1. The old fixed points exist only when dim = dim T ; they are all the connected components Fi of MT for which µ (Fi ) is in the interior of . The set of T fixed points at zero is defined to be the connected component µ−1 (0) of M , which is just the symplectic reduction M0 . The new fixed points are all the other connected components Fi of MT . It is not difficult to see that every Fi is also a connected component of the fixed point set M T , while Fi do not correspond to any fixed points on M. 2.3 Kirwan map We recall the definition of equivariant cohomology HT∗ (M) with complex coefficients using the Cartan model. Denote

∗T (M) = S(t∗ ) ⊗ ∗ (M)T , where S(t∗ ) denotes the algebra of polynomials on t and ∗ (M)T denotes all T invariant differential forms. So, if f ∈ S(t∗ ), α ∈ ∗ (M)T and X ∈ g we set (f ⊗ α)(X) = f (X)α. The T -equivariant differential on ∗T (M) which defines the equivariant cohomology is given by dT (f ⊗ α) = f ⊗ dα − xi f ⊗ ıξ i α, M

i is the vector where ξ1 , . . . , ξd is a basis of g; x1 , . . . , xd is the dual basis of t∗ ; and ξM ∗ i field generated by the action of ξ . If the equivariant form β ∈ T (M) is closed, that is dT β = 0, we denote by [β] the cohomology class it represents. If T acts locally freely on M, then it is well known that

HT∗ (M) = H ∗ (M/T ), and if the action is trivial, then HT∗ (M) = H ∗ (M) ⊗ S(t∗ ) = H ∗ (M) ⊗ HT∗ (pt).

Localization theorems by symplectic cuts

309

For p ∈ t∗ let ip be the inclusion µ−1 (p) → M. If p is a regular value of the moment map, then T acts locally freely on µ−1 (p) so that HT∗ (µ−1 (p)) ∼ = H ∗ (µ−1 (p)/T ) = H ∗ (M//p T ).

(2.1)

Composition of the pullback ip∗ with the isomorphism (2.1) defines the Kirwan map κp : HT∗ (M) → H ∗ (M//p T ). Kirwan [K] showed that if M is compact this map is surjective. In the presence of another Hamiltonian action on M by a torus T which commutes with the action of T , the Kirwan map generalizes to its equivariant version: κp : HT∗×T (M) → HT∗ (M//p T ). Kirwan surjectivity was generalized to this case in [Go]. Analogously, in the case when T = H × S and p ∈ µ(M H ) we can define the Kirwan map κpH : HS∗ (M H ) → H ∗ (M H //p S). We will mostly be interested in the equivariant version of this map. Let us take account of the trivial action of H on both M H and M H //p S. So in the rest of the paper κpH will be the map κpH : HT∗ (M H ) → HH∗ (M H //p S). (2.2) Let us now apply the equivariant version of the Kirwan map to symplectic cuts with respect to cones. Given a cone = β , the product T × T acts on M × Cβ and the symplectic cut M is produced by reducing M × Cβ at 0 with respect to the T action. So if we think of T × T as the product of T × e and T , then the equivariant version of the Kirwan map produces the map κ : HT∗×T (M × Cβ ) → HT∗×e (M ) = HT∗ (M ). As mentioned before, the action of T on M might not be effective, since the torus T orthogonal to the cone acts trivially on M . In particular, HT∗ (M ) = HT∗/T (M ) ⊗ HT∗ (pt). For η ∈ HT∗ (M) denote by η the class κ (η ⊗ 1) ∈ HT∗ (M ). It is an easy exercise to see that η ∈ HT∗/T (M ) ⊗ 1. Let us also notice that if Fi is a connected component of the fixed point set of both M and M with µ(Fi ) = µ (Fi ) ∈ Int(), then ι∗Fi η = ι∗Fi η , where by abuse of notation we denote by ιFi both the inclusion of Fi into M and into M . (Because is transverse to µ(M), the existence of such Fi implies that the dimension of the cone is at least the dimension of µ(M).) It is also easy to see that ιM0 η = κ0 (η) ⊗ 1 ∈ H ∗ (M0 ) ⊗ 1 ⊂ HT∗ (M0 ),

(2.3)

where, since T acts trivially on M0 , we know that HT∗ (M0 ) = H ∗ (M0 ) ⊗ S(t∗ ).

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2.4 ABBV localization theorem Suppose that M is compact, oriented and carries the action of a torus T . The pushfor ward map from HT∗ (M) to HT∗ (pt) is the integration over M and is denoted by . The theorem of Atiyah–Bott and Berline–Vergne (or just the ABBV theorem) [AB, BV] states that for η ∈ HT∗ (M) η= M

Fi

ι∗Fi (η) Fi

e(ν(Fi ))

.

(2.4)

Here Fi are the connected components of the fixed point set M T , ιFi : Fi → M are their inclusions, ν(Fi ) are the normal bundles of Fi , and e(ν(Fi )) are their T equivariant Euler classes. We need to know more about these T -equivariant Euler classes. Because of the splitting principle [BT] we can assume without loss of generality that e(ν(Fi )) splits as a sum of line bundles L1 ⊗ · · · ⊗ Lk . Assume T acts on the fibers of Li with weight λi . Then the T -equivariant Euler class is 1 (λi + c1 (Li )), (2.5) e(ν(Fi )) = where c1 (Li ) is the first Chern class of Li . TheABBV localization formula was generalized to orbifolds by Meinrenken [Me]. We refer to [Me] for details. Let us just mention that the only difference with (2.4) is the appearance of constants before each term of the formula: 1 ι∗Fi (η) 1 η= , (2.6) dM M dFi Fi e(ν(Fi )) Fi

where for a connected orbifold X, the size of the finite stabilizer at a generic point of X is equal to dX . Moreover (2.5) is still a valid formula for orbifolds, where the λi (when properly interpreted) are rational weights of the action on the normal bundle. Another important property of the equivariant Euler classes is the following generalization of [GK, Proposition 3.1]. Proposition 2.2. Assume T = S × H , π : t∗ → s∗ is the natural projection, p ∈ µ(M H ), and q = π(p). Then κpH : HT∗ (M H ) → HH∗ (M H //p S) takes the T -equivariant Euler class of the normal bundle of M H onto the H -equivariant Euler class of the normal bundle of M H //p S in M//q S. Proof. The argument is almost identical to the one used in [GK]. Namely, let Z = µ−1 (p) ∩ M H and let ρ be the projection from Z to M H //p S and i : Z → M H . Then i ∗ ν(M H ) = ρ ∗ ν(M H //p S). The proposition follows from functoriality of the Euler class as a map from oriented vector bundles to cohomology.


311

3 Residues In this section we define the residue operations and discuss their basic properties. Most of the definitions and results of this section have appeared before in either [JK1] or [JK2]. However, we repeat all the definitions of different kinds of residues (equations (3.1), (3.2), (3.8), (3.11), (3.12), (3.15), and (3.16)), so that these definitions can be understood without referring to the above sources. At the same time, for shortness, we do not repeat the arguments of [JK1] or [JK2], which prove the significance of these definitions, and do not repeat the proofs of certain properties of residues. 3.1 Residues of meromorphic 1-forms in one variable Think of the Riemann sphere as the one point compactification C∪{∞} with the complex coordinate z on C. Let f (z) be a meromorphic function on the Riemann sphere with values in a topological vector space V which can be written as the finite sum f (z) = gj (z)eiλj z , j

where gj (z) are rational functions of z and λj ∈ R. Then in the case when all λj = 0 we define Res(f dz) = res(gj (z)eiλj z ; z = b) (3.1) λj >0 b∈C

as was done in [JK2]. The other case we will be interested in is when λj = 0 for all j ; then we define Res(f dz) = lim Res(f (z)eisλz dz) (3.2) s→0+

for some λ > 0. It is easy to see that in this case Res(f dz) is just the sum of all residues on C and since the sum of all residues of a meromorphic function is zero we conclude that Res(f dz) = −resz=∞ (f dz). Given a linear map ψ : V → W between two topological spaces, the residue commutes with it ψ(Res(f )dz) = Res(ψ(f )dz). (3.3) In the case when V carries an algebra structure, an example which will be important for us is the residue of the function of the form f =

g(z) , cz + a

where a ∈ V , c ∈ C − {0}, and g(z) is a polynomial in z with values on V . For A = az use 1 = 1 − A + A2 − . . . , (3.4) 1+A 0 a j to rewrite f as a sum m j =−∞ γj z for γj ∈ V , which converges for | z | < 1.

312


Let w =

1 z

be another coordinate on the Riemann sphere. Then ∞

γ−j w j

j =−m0

−dw w2

is the Taylor expansion of f dz at w = 0. Hence ⎛ ⎛ ⎞ ⎞ m0 ∞ γj zj dz⎠ = resw=0 ⎝ γ−j w j −2 dw⎠ = γ−1 . Res(f dz) = −resz=∞ ⎝ j =−∞

j =−m0

(3.5) In the case when g(z) is just a constant g0 ∈ V , we get Res(f dz) =

g0 . c

(3.6)

We emphasize that the residue is well defined only as a function of meromorphic 1-forms, not functions; the residue at 0 of the 1-form f (z)dz is independent of the choice of coordinate z. (The residue is invariant under a change of variables z → g(z) provided that g(z) is a meromorphic function of z and dg(0) = 0, whereas this is not true of usual definition of the residue at 0 of a meromorphic function.) 3.2 Residues of functions of several variables Let us now consider a function f of several complex variables with values in a topological space V . More precisely, we assume f is defined on the complexified Lie algebra tC = t ⊗ C of the torus T , and f is a linear combination of functions of the form q(X)eiλ(X) h(X) = 8k (3.7) j =1 αj (X) for some polynomials q(X) of X ∈ tC , with values in V , λ ∈ t∗ and some α1 , . . . , αk ∈ t∗ − {0}. Choose a coordinate system X1 , . . . , Xm on t, and denote by the same letters the complexified coordinates which provide a coordinate system of tC . Let t be the subspace of t given by zeros of X1 , . . . , X . Define Resm (hdXm ) = Res(hdXm ),

(3.8)

where the variables X1 , . . . , Xm−1 are held constant while calculating this residue. As explained in [JK2, Remark 3.5(1)], in the case λ = 0 the residue Resm is well defined only for a generic choice of coordinates X1 , . . . , Xm (the precise condition on the coordinates being specified in this remark). Moreover, by [JK2, Remark 3.5(2)], Resm (f dXm ) is a linear combination of functions of the form iλ(X) q(X)e ˜ ˜ h(X) = 8k−1 , ˜ j (X) j =1 α

(3.9)


313

where q(X) ˜ is a polynomial on the complexification of t/tm−1 and α˜ j are in the dual of t/tm−1 . To consider the case when λ = 0, in other words h0 (X) = 8k

q(X)

(3.10)

,

j =1 αj (X)

we may make a choice of λ0 ∈ t∗ for which λ0 (X) = define Resm (h0 dXm ) as

m

0 j =1 λj Xj

with λ0m > 0 and

0

Resm (h0 dXm ) = lim Resm (h0 eisλ dXm ).

(3.11)

s→0+

We can easily check that the residue Resm is a continuous function of s ∈ R+ and this limit exists, so we can define Resm (hdXm ) even when λ = 0. It is still true in this situation that Resm (f dXm ) is a linear combination of functions of the form given in (3.10) with λ = 0. In the case when V is an algebra, an important generalization of (3.6) is the following.

Lemma 3.1. Resm

g0 dXm c i i Xi + v

=

g0 , cm

where g0 , v ∈ V and ci ∈ C. Proof. The proof follows from (3.5) after setting c = cm and a = + v.

m−1 i=1

ci Xi

3.3 Iterated residues We again consider functions f which are linear combinations of functions of the form (3.7). As was just explained, Resm (f dXm ) is a linear combination of functions of the form (3.9), which allows us to take the residue of this function again. So we set Resm m = Resm and by induction define the iterated residue m m m Resm (f [dX] ) = Res(Res+1 (f [dX]+1 )dX ),

(3.12)

where [dX]m stands for the form dX ∧ · · · ∧ dXm and, as above, the coordinates m X1 , . . . , X−1 are held constant while calculating this residue. Clearly Resm (f [dX] ) is a function on the complexification of t/t−1 . In the case V is an algebra, a generalization of Lemma 3.1 states the following. Lemma 3.2. For a generic choice of coordinates X1 , . . . , Xm , ' * g0 g 0 Resm = , [dX]m 8m−+1 det( α) ˜ (αi (X) + vi ) i=1 where g0 , vi ∈ V , αi ∈ t∗ −{0}, and α˜ is the the matrix {aij }1≤i≤m−+1;≤j ≤m , where αi (X) = aij Xj .

314


Proof. The proof is analogous to the proof of property (iv) for the iterated residue in [JK2, Proposition 3.4]. Notice that for h0 defined in (3.10) the definition of m ) is given in [JK2] as the limit as s → 0+ of Resm (h0 eisλ(X) [dX]m ) 0 Resm (h [dX] where λ(X) = j λj Xj and we choose λ so that all the λj satisfy λj > 0.

Given a linear map ψ : V → W between two topological spaces, the iterated residue commutes with this map: m m m ψ(Resm (f [dX] )) = Res (ψ(f )[dX] ).

(3.13)

3.4 Residues with respect to cones Iterated residues depend on the choice of coordinates on t. Fix an inner product on t. Let us define residues which depend only on this inner product and a choice of a certain cone in t. We introduce a function f which is a linear combination of functions of the form (3.7). We consider the set where none of the functions αj appearing in the denominators of functions h become zero, namely the set {X ∈ t : αj (X) = 0 for all αj }.

(3.14)

Let be an open cone which is a connected component of this set. Then for a generic choice of coordinate system X = (X1 , . . . , Xm ) on tC for which (0, . . . , 0, 1) ∈ define the residue with respect to the cone by Res (h[dX]) = /Resm 1 (h[dX]),

(3.15)

[dX]m 1

where [dX] = and / is the determinant of any (m) × (m) matrix whose columns are the coordinates of an orthonormal basis of t defining the same orientation on t as the chosen coordinate system. To guarantee that Res (h[dX]) is well defined (where h is of the form (3.7)), we need to make one additional assumption: we assume that λ is not in any proper subspace of t spanned by some αi ’s. It was shown in [JK2] that under the above assumptions Res (h[dX]) is well defined, does not depend on the choice of the coordinates but only on the choice of the cone and the inner product on t. Originally, the residue Res was introduced in [JK1] as a generalization of a certain integral over a vector space. In [JK2, Proposition 3.4], it was shown that the definition (3.15) coincides with the original definition of Res from [JK1]. In [JK2, Proposition 3.2] it was shown that certain properties together with linearity uniquely define Res . Let us recall these properties: 1. Let α1 , . . . , αv ∈ ∗ be vectors in the dual cone. Suppose that λ is not in any cone of dimension m − 1 or less spanned by a subset of the {αi }. If J = (j1 , . . . , jm ) j j is a multiindex and XJ = X11 . . . Xmm , then ' * J iλ(X) [dX] X8e =0 Res v i=1 αi (X) unless all of the following properties are satisfied:


315

a) {αi }vi=1 span t∗ as a vector space, b) v − (j1 + · · · + jm ) ≥ m, c) λ ∈ α1 , . . . , αv + , the positive span of the vectors {αi }. 2. If properties (1)(a)–(c) above are satisfied, then ' ' * * J iλ(X) [dX] J k eisλ(X) [dX] X8e X (iλ(X)) 8 Res = , lim Res v k! vi=1 αi (X) s→0+ i=1 αi (X) k≥0

and all but one term in this sum are 0 (the nonvanishing term being that with k = v − (j1 + · · · + jm ) − m). 3. The residue is not identically 0. If properties (1)(a)–(c) are satisfied with α1 , . . . , αm linearly independent in t∗ , then ' * iλ(X) [dX] e 1 Res 8m , = det(α) α (X) i=1 i where α is the nonsingular matrix whose columns are the coordinates of α1 , . . . , αm with respect to any orthonormal basis of t defining the same orientation. When λ is of the form ki=1 si αi , where fewer than m of the si are nonzero, then we define ' ' * * i(λ(X)+sρ(X)) [dX] eiλ(X) [dX] 8 e 8 = lim Res , (3.16) Res v v s→0+ i=1 αi (X) i=m αi (X) where ρ ∈ t∗ is chosen so that ρ(ξ ) > 0 for all ξ ∈ , and for small s, λ + sρ does not lie in any cone of dimension m − 1 or less spanned by a subset of the {βj }. We will need another property of residues. Lemma 3.3. Let f (X1 , . . . , Xm ) be a function on t given by a linear combination of functions of the form (3.7) with λ = 0. Moreover, assume that for every set of values a1 , . . . , am−1 of the variables X1 , . . . , Xm−1 the function g(z) = f (a1 , . . . , am−1 , z) is holomorphic. Let be an appropriate choice of cone such that Res (f [dX]) is defined, in particular contains the point (0, . . . , 0, 1). Then Res (f [dX]) = Res− (f [dY ]), where Y1 , . . . , Ym is a set of coordinates such that (0, . . . , 0, 1) ∈ −. Proof. For fixed a1 , . . . , am−1 , let g(z) =

gj (z)eiλj z .

Then Res(g(z)dz) = res+ (g(z)dz) =

λj >0 b∈C

res(gj (z)eiλj z ; z = b).

(3.17)

316


Define

res− (g(z)dz) =

res(gj (z)eiλj z ; z = b).

λj 1, then in terms of the same notation Gi are the new fixed points.) Recall that any equivariant cohomology class η ∈ HT∗ (M) descends to a class η on M : η = κ (η ⊗ 1) ∈ HT∗/T (M ) ⊗ 1 ⊂ HT∗ (M ).


317

Think of η as a class in HT∗/T (M ) and apply the orbifold version of the ABBV localization theorem to it: 1 ι∗G (η ) 1 κ0 (η) 1 i + , (4.1) η = dM M dM0 M0 e(ν(M0 )) dGi Gi e(ν(Gi )) Gi

where ιGi are the inclusions of Gi into M and the Kirwan map at zero κ0 appears because of (2.3). Apply the residue operation to both sides of (4.1). For this we have to specify a coordinate X1 on the one-dimensional Lie algebra of T /T . Clearly the dual of this Lie algebra can be identified with the line in t∗ passing through the cone . So β defines a coordinate on the Lie algebra of T /T , and we define Xβ = X1 to be this coordinate. Using X1 we get the formula ι∗ (η ) dXβ dXβ dXβ κ0 (η) Gi Res1 + . η = Res1 Res1 dM M dM0 M0 e(ν(M0 )) dGi Gi e(ν(Gi )) Gi

(4.2) Since M η is just a polynomial function on the Lie algebra of T /T , by (3.5) the left-hand side of (4.2) is zero. The normal bundle ν(M0 ) is just a line bundle whose equivariant Euler class is given by e(ν(M0 )) = Xβ + c1 (ν(M0 )), (4.3) where c1 (ν(M0 )) is the first Chern class of ν(M0 ). Thus by (3.13) and (3.6) dXβ κ0 (η)dXβ κ0 (η) 1 Res1 =(††) Res1 dM0 M0 e(ν(M0 )) dM0 M0 Xβ + c1 (ν(M0 )) 1 = κ0 (η). dM0 M0 κ0 (η) Remark 4.1. To show that (††) follows from (3.13) think of e(ν(M as a function on 0 )) ∗ ∗ t with values in H (M). If we define ψ : H (M) → C to be the usual integration on M, then (3.13) applied to this ψ yields (††).

Hence (4.2) yields a formula for the integral of κ0 (η) over M0 of the Kirwan map of η in terms of the residues of certain integrals over the Gi . To put this formula in the form in which it appeared in [GK] let us transform the terms corresponding to the Gi in (4.2) by commuting Res1 with the integration and the Kirwan map. By (3.13) and Proposition 2.2, we have ' ' ' ∗ * * ι∗ (η ) * ιMi η dXβ 1 Gi Hi Res1 = dXβ , Res1 κpi dGi Gi e(ν(Gi )) dGi Gi e(ν(Mi )) where ιMi is just the inclusion of Mi into M, and as defined in (2.2) κpHii is the Kirwan map from HT∗ (Mi ) to HT∗/T (Gi ).

318


Notice that each Mi is fixed by the one-dimensional torus Hi , so that the Lie i on t such that algebra hi is a subspace of t. Pick a coordinate system X1i , . . . , Xm i i i Xm = β and X1 , . . . , Xm−1 vanish on hi , so that tm−1 = hi . Then it is not difficult to see that Res1 ◦ κpHii = κpHii ◦ Resm,i , where Resm,i is Resm defined using the coordinate system {Xji } (note that the definition of Resm was given in (3.11)). This allows us to obtain the following restatement of [GK, Theorem 3.1]. Theorem B. For η ∈ HT∗ (M) κ0 (η) = − M0

'

dM 0

Gi

dGi

Gi

κpHii Resm,i

ι∗Mi η e(ν(Mi ))

* dβ .

(4.4)

Guillemin and Kalkman iterated this result using certain combinatorial objects called dendrites to produce a formula for M0 κ0 (η) in terms of the integration over the connected components of the fixed point set M T of the original T action on M. We will discuss dendrites and their generalizations in Section 4.3. 4.2 Higher-dimensional generalization of Guillemin–Kalkman localization We now generalize the formula of the previous section to the case when we cut with a cone of any dimension. As before, let (M, ω) be a compact symplectic manifold with an effective Hamiltonian T action. Let µ : M → t∗ be the moment map. Pick any cone transverse to µ. Assume is generated by the linearly independent weights β1 , . . . , βk . Recall that in Definition 2.1 we distinguished three kinds of fixed points of M : the old fixed points (whose connected components are denoted by Fi ), the new fixed points (whose connected components are denoted by Fi ), and the symplectic reduction M0 . As in the case of one-dimensional cones any equivariant cohomology class η ∈ HT∗ (M) descends to a class η on M η = κ (η ⊗ 1) ∈ HT∗/T (M ) ⊗ 1 ⊂ HT∗ (M ). As before, we think of η as a class in HT∗/T (M ) and apply the ABBV localization theorem to it: 1 ι∗F (η ) κ0 (η) 1 1 i + η = dM M dM0 M0 e(ν(M0 )) dFi Fi e(ν(Fi )) Fi (4.5) ∗ 1 ιF (η ) i + . dFi Fi e(ν(Fi )) Fi

Here, κ0 is the Kirwan map at zero and ιFi , ιFi are the inclusions of Fi , Fi into M .


319

Let us apply the iterated residue operation to both sides of (4.5). As in the onedimensional case the dual of the Lie algebra of T /T can be identified with the subspace in t∗ passing through the cone . Consider the set of weights {αi } which appear in the isotropy representation of the T /T action at the connected components of the fixed point set of the T /T action on M . Notice that the weights β˜1 , . . . , β˜k of the isotropy representation of T /T at M0 are the images of the weights β1 , . . . , βk under the map (t/t )∗ → t∗ . In particular, the set {αi } contains the weights β˜i . Let {X1 , . . . , Xk } be a generic coordinate system on T /T such that the determinant of the matrix which expresses β˜i as a linear combination of Xj is one. Then by applying Resk1 to both sides of (4.5) we get the formula 0=

[dX]k1 Resk1 dM0

M0

[dX]k1 κ0 (η) + Resk1 e(ν(M0 )) dFi

Fi

+

Fi

[dX]k1 Resk1 dFi

ι∗Fi (η ) Fi

e(ν(Fi )) ι∗F (η ) i

Fi

e(ν(Fi ))

(4.6) ,

where the left-hand side is zero since M η is just a polynomial function on the Lie algebra of T /T . The weights of the isotropy representation of T /T on the normal bundle ν(M0 ) are just β˜i . Hence ν(M0 ) splits as a direct sum of line bundles ⊕i Li , where T /T acts on the fibers of Li by the weights β˜i . Then the Euler class of ν(M0 ) is 1 (β˜i + c1 (Li )), (4.7) e(ν(M0 )) = i

where c1 (Li ) are the first Chern classes of Li . Thus by (3.13) (see also Remark 4.1) and Lemma 3.2, we have [dX]k1 1 κ0 (η) = κ0 (η). (4.8) Resk1 dM0 M0 e(ν(M0 )) dM0 M0 By analogy with the one-dimensional case, we should now simplify the second and third terms of the right-hand side of (4.6). But the second term is already in the form we want since it is written in terms of the fixed points of M. To simplify the last term of (4.6), first consider the situation when a point pi = µ (Fi ) is an intersection of the interior of with a wall of µ(M) of dimension r > 0. Assume that this wall is the moment map image of Mi , which is stabilized by Hi ⊂ T . Then by (3.13) and Proposition 2.2, we have ' ' ' ∗ ** ι∗ (η ) * ιMi η 1 1 Fi k k k k Hi = Res1 [dX]1 Res1 [dX]1 κp , i dFi dFi Fi e(ν(Mi )) Fi e(ν(Fi )) (4.9) where ιMi is just the inclusion of Mi into M, and as defined before κpH i is the Kirwan map from HT∗ (Mi ) to HT∗/T (Fi ).

i

320


For the more general situation when pi is an intersection of any face of with a wall of µ(M) of complementary dimension, formula (4.9) becomes a little more complicated. Namely the Euler class of Fi is no longer a Kirwan map image of the Euler class of Mi , but rather this is multiplied by another class νi . The class νi can be understood as follows. Take the symplectic cut M,i of Mi with respect to the cone . This symplectic cut sits naturally inside M . Then νi is the Euler class of the normal bundle of Fi inside M,i . While this class can be quite complicated, by the generalized Kirwan surjectivity theorem of [Go] we know that there exists a class τi on Mi such that κpH i (τi ) = νi . So we conclude that i

'

1 Resk1 [dX]k1 dFi

ι∗F (η )

*

i

Fi

e(ν(Fi ))

1 = dFi

'

Fi

Resk1

'

[dX]k1 κpH i i

ι∗Mi η e(ν(Mi ))τi

** .

i } To simplify this term even further, let us choose a set of coordinates {X1i , . . . , Xm on t as follows. Each Mi is fixed by a subtorus Hi of T , so that its Lie algebra hi lies inside t. (Notice that dim Hi ≤ dim and this inequality might be strict.). i Choose any generic coordinates X1i , . . . Xm−k which vanish on hi and coordinates i i Xm−k+1 , . . . , Xm , which are the images of X1 , . . . , Xk under the map (t/t )∗ → t∗ . Then we conclude that

Resk1 ◦ κpH i = κpH i ◦ Resm m−k+1 , i

i

i i where Resm m−k+1 on the right-hand side is taken with respect to coordinates X1 , . . . , Xm . Thus we get the following generalization of [GK, Theorem 3.1] to the case of cones of arbitrary dimension.

Theorem C. For η ∈ HT∗ (M), κ0 (η) = − M0

dM 0

Fi

−

dFi

dM

Fi

0

Fi

dFi

Fi

Resk1 [dX]k1

ι∗Fi (η ) e(ν(Fi ))

i m κpH i Resm m−k+1 [dX ]m−k+1 i

ι∗Mi η e(ν(Mi ))τi

(4.10) .

4.3 Dendrites and their generalizations In addition to Theorem B, Guillemin and Kalkman [GK] proved a formula which uses Theorem B iteratively to express M0 κ0 (η) in terms of integration over the connected components of M T . They used the term “dendrites’’ to designate the combinatorial objects responsible for how the iteration is performed. Consider a finite collection D of tuples ((q), W ), where (q) is a onedimensional shifted cone (that is, if ⊂ t∗ is a cone centered at the origin and q ∈ t∗ , then (q) = {x + q | x ∈ }) and W is a wall of µ(M) such that (q) lies inside the affine space spanned by W . Notice that according to our conventions


321

every W uniquely defines a subtorus HW of T and a connected component MW of M HW such that W = µ(MW ).) Assume that D contains a tuple (0 (0), µ(M)) (we will treat 0 as the cone used in Theorem B). Then we say that D is a dendrite if the following conditions hold: 1. For ((q), W ) ∈ D, the cone (q) is transverse to µ(MW ), 2. For ((q), W ) ∈ D, if (q) intersects a codimension one wall W of µ(MW ) at a point q , then there is a unique cone such that ( (q ), W ) ∈ D. Obviously it is possible to construct a dendrite which contains a tuple (0 (0), µ(M)) as long as 0 is transverse to µ(M). Now consider formula (4.4) of Theorem B produced using the cone 0 . Assume we are given a dendrite D containing (0 (0), µ(M)). Every term in the summation on the right-hand side of (4.4) corresponds to an intersection pi = µ (Gi ) of 0 with a codimension one wall Wi . By definition of the dendrite, there exists a unique cone i such that (i (pi ), Wi ) ∈ D. Set Hi = HWi and Mi = MWi and notice that Gi = Mi //pi (T /Hi ). Moreover, let us shift the moment map on Mi by defining µi = µ − pi . Then, we can apply Theorem B to the T /Hi action on Mi and the cone i to compute ' * ι∗Mi η Hi κpi Resm dXm e(ν(Mi )) Mi //p (T /Hi ) i

as a sum of integrals over symplectic reductions of the form N //(T /H ), where H is a two-dimensional subtorus of T and N isa connected component of M H . Repeating this process we can express M0 κ0 (η) as a summation of integrals over the connected components of the fixed point set M T . More specifically, for a dendrite D we say that the sequence of tuples from D ((0 (q0 ), W0 ), (1 (q1 ), W1 ), . . . , (k (qk ), Wk )) is a path P if (0 , µ(M)) = (0 (q0 ), W0 ); Wk is zero-dimensional, so that there is a connected component F of M T with µ(F ) = Wk (we will denote this F by FP ); each qj is an intersection of j −1 (qj −1 ) with a codimension one wall Wj of µ(MWj −1 ). For a path P , let kj = dim Wj . Then for γ ∈ HT∗/HW (MWj −1 ) and an appropriately j −1

chosen set of coordinates on the Lie algebra of T /HWj −1 define ' * ι∗MW γ j Qj (γ ) = −Reskj dXkj . e(ν(MWj )) For a path P , define QP = Qk ◦ · · · ◦ Q1 . The above discussion proves the following. Theorem D. For a dendrite D and η ∈ HT∗ (M), κ0 (η) = dM0 QP (η), M0

P

FP

322


where the above sum is taken over all possible paths in D. Now consider a collection D of tuples ((q), W ), where (q) is a shifted cone of any dimension and W is a wall of µ(M) such that (q) lies inside the affine space spanned by W . Again, every W uniquely determines a subtorus HW of T and a connected component MW of M HW such that W = µ(MW ). Assume that D contains a tuple (0 (0), µ(M)). Then we say that D is a multidimensional dendrite if the following conditions hold 1. For ((q), W ) ∈ D the cone (q) is transverse to µ(MW ), 2. For ((q), W ) ∈ D if a face of (q) of dimension r ≤ dim W intersects a wall W of µ(MW ) of dimension dim W − r at a point q , then there is a unique cone such that ( (q ), W ) ∈ D. In analogy with the case of dendrites of one-dimensional cones, consider formula (4.10) of Theorem C produced using the cone 0 . Assume we are given a multidimensional dendrite D containing (0 (0), µ(M)). Every term in the second summation on the right-hand side of (4.10) corresponds to a new connected component Fi of MT . Moreover, its moment map image pi = µ (Fi ) is always an intersection of a face of with a wall Wi of complementary dimension. By definition of the multidimensional dendrite, there exists a unique cone i such that (i (pi ), Wi ) ∈ D. (Notice that MWi and HWi are just Mi and Hi in the notation of Theorem C.) As in the case of one-dimensional cones, we know that Fi = Mi //pi (T /Hi ), so we can apply Theorem C to the T /Hi action on Wi and the cone i (pi ) to compute ' * ι∗Mi η Hi m i m κp Resm−k+1 [dX ]m−k+1 i e(ν(Mi ))τi Mi //p (T /Hi ) i

as a sum of integrals over symplectic reductions of the form N //(T /H ), where H is a subtorus of T of dimension at least 2 and N is a connected component of M H . Using the multidimensional dendrite we can iterate the process and express T M0 κ0 (η) as a summation of integrals over the connected components of M as follows. For a multidimensional dendrite D we say that the sequence of tuples ((0 (q0 ), W0 ), (1 (q1 ), W1 ), . . . , (k (qk ), Wk )) is a path P if (0 , µ(M)) = (0 (q0 ), W0 ); Wk is zero-dimensional, so that there exists a connected component F of M T with µ(F ) = Wk (again we denote FP = F ); each qj is the intersection of the interior of a face σ of j −1 (qj −1 ) with a wall Wj of µ(MWj −1 ) such that dim σ + dim Wj = dim Wj −1 . For a path P , let kj = dim Wj and mj = dim j . Then for γ ∈ HT∗/HW (MWj −1 ) and an appropriately chosen set j −1

of coordinates on the Lie algebra of T /HWj −1 define ' Qj (γ ) = For a path P define

k −Reskjj −mj +1

* ι∗MW γ kj j [dX]kj −mj +1 . e(ν(MWj ))


323

QP = Qk ◦ · · · ◦ Q1 . It is clear that Theorem D holds in the case when D is a multidimensional dendrite.

5 New proof of the Jeffrey–Kirwan localization formula As explained in the previous section, it is possible to iterate the formulas of Theorems B and C using (multidimensional) dendrites to express integration of κ0 (η) over M0 as a sum of integrals of certain forms over the connected components of M T . In this section we present another way of writing such a formula. The rough idea is to choose a very wide cone , whose dual is inside a certain cone , then apply the residue operation with respect to to the ABBV formula for ηei ω˜ (where ω˜ is the equivariant symplectic form) in such a way that the terms corresponding to the new fixed points Fi of M are zero. As a result we will obtain a new proof of the Jeffrey–Kirwan localization theorem [JK1]. 5.1 Choice of the cone In this section we explain how to choose the cone . It is convenient to think of as a very wide cone, in other words a cone whose boundary is close to being a hyperplane. Given an effective Hamiltonian action of T on a compact manifold M, let {αi } be the set of all weights appearing in the isotropy representation of T at the fixed points. Pick a connected component of the set {ξ ∈ t|αi (ξ ) = 0 for all i}. Consider the dual cone ∗ = {X ∈ t∗ |X(ξ ) ≥ 0 for all ξ ∈ }. Now pick a cone transverse to µ(M) spanned by m = dim t weights β1 , . . . , βm such that satisfies 1. ∗ ⊆ , or in other words ∗ ⊆ , 2. For every wall W of µ(M), if W ∩ is not empty, then there exists ξW ∈ ∗ such that the maximum of q(ξW ) for q ∈ W ∩ is attained at a vertex of W . Let us explain why such a cone always exists. Pick a rational vector ξ0 ∈ and let H be the hyperplane in t∗ annihilated by ξ0 . For a weight p in the interior of ∗ define Hp = H + p. Then Hp ∩ ∗ is a rational polytope. In particular, there exists a simplex S ⊂ Hp with rational vertices β˜1 , . . . , β˜m which contains the polytope Hp ∩ ∗ . Take the weights β1 , . . . , βm , which define , to be multiples of β˜1 , . . . , β˜m . Clearly satisfies (1). Moreover, by increasing the size of S, that is by making wider, we can always guarantee that satisfies (2). Since there are infinitely many choices of simplices S, there is a choice of S for which is transverse to µ(M). Now consider the symplectic cut M and the set {γi } of all the weights which appear as weights of isotropy representations at fixed points of M . Consider the set ∗ ∩ {ξ ∈ t|γi (ξ ) = 0 for all i},

324


¯ be a connected component of this set. and let the cone For each connected component F of MT , let {γjF } be the set of weights of the ¯ that is if isotropy representation of T at F . Polarize the weights {γjF } using , F F F F F ¯ γj (ξ ) < 0 for all ξ ∈ then set γ¯j = γj , otherwise let γ¯j = −γj . Define CF to be the cone containing all the points of the form µ (F ) + sj γ¯jF with sj being nonnegative real numbers. If F is an old connected component of the fixed point set, then the polarization ¯ is the same as using , since ¯ ⊂ . If F = M0 , then of the weights {γjF } using CF = −. For the new fixed points let us prove the following important fact. Lemma 5.1. Let F be a new connected component of the fixed point set MT . Then the cone CF does not intersect the interior of . Proof. Let p = µ (F ). Since intersects µ(M) transversely, there is a subtorus H of T and a connected component M of M H for which F is the symplectic reduction of M at p. Moreover, p is just the intersection of the wall W = µ(M ) of dimension k and an open face σ of of dimension m − k. Let us order the weights {γjF }nj=1 of the isotropy representation of T at F in a special way. Assume that each of the first k weights is parallel to an intersection W ∩ σ , where σ is an open face of such that dim σ = dim σ + 1 and the closure of σ contains σ . Assume also that each of the last n − k weights is parallel to an intersection W ∩ σ , where W is a wall with dim W = dim W + 1 and W ⊂ W . (It is easy to see that every γjF falls into one of these categories.) Let CF1 be the cone spanned by the first k polarized weights centered at the origin and let CF2 be the cone spanned by the other weights, also centered at the origin. Then CF = p + CF1 + CF2 . Since the cone p + CF2 lies in the affine space passing through σ , it remains to show that p + CF1 does not intersect the interior of . If two of the weights γjF are parallel, then we can remove one of them without changing the polarized cone F . Since the first k weights point in exactly k different directions (there are precisely k faces σ of with σ ⊂ σ¯ and dim σ = dim σ + 1), we can assume without loss of generality that k = k. Let the first k weights span a cone C˜ F centered at the origin. It is clear that in a small neighborhood of p the polytope ∩ W is equal to the cone p + C˜ F . Moreover, since the first k weights are linearly independent, the cones C˜ F and CF1 are either the same or do not have common points in the interior. So it remains to show that C˜ F and CF1 are different, which is the same as showing that during polarization at least one of the first k weights changes sign. So, we must show that it is impossible to have γjF (ξ ) < 0 for 1 ≤ j ≤ k for ¯ If this happens then the maximum of q(ξ ) for q ∈ W ∩ is attained at every ξ ∈ . µ (F ), which is impossible, by property (2) of the cone .

5.2 Jeffrey–Kirwan localization ¯ and be defined as in the previous section. Consider the symplectic Let cones , cut M . Let p ∈ be a point close to the origin. Then µε = µ − εp for ε > 0 is


325

a moment map on M . Define ω˜ ε = ω + iµε to be an equivariant symplectic form on M , where ω is the symplectic form on M . For a form η ∈ HT∗ (M), there corresponds a form η ∈ HT∗ (M ). Apply the ABBV localization theorem to get ε η eω˜ ε = IM + IFεi + IFε , (5.1) 0 i

M

where for F = M0 , Fi , or Fi , ∗ ∗ ιF (η eω ) ιF (η eω ) 1 i(µ (F )−εp) 1 i(µε (F )) = . e e IFε = dF dF F e(ν(F )) F e(ν(F )) ¯ and −: ¯ Let us now apply Lemma 3.3 to the function M η eω˜ ε and cones ¯

¯ η eω˜ ε ) = Res− [dX]

Res ([dX] M

η eω˜ ε . M

Hence by (5.1) we get

¯ ε ε + I + IFε Res [dX] IM Fi 0 i

¯ − ε ε = Res I Fi + IFε . [dX] IM0 +

(5.2)

i

Let us show that four of the six terms of (5.2) are zero. Indeed by Lemma 5.1 the cones CFi do not contain εp. Hence by property (1) of the residue, we get ¯ Res (IFε ) = 0. i

Analogously, since the cone CM0 does not contain εp ¯

ε Res (IM ) = 0. 0

Similarly, for small enough ε the cones −CFi and −CFj do not contain εp. Hence by property (1) of the residue, we have ¯

Res− (IFε ) = 0, i

¯

Res− (IFεj ) = 0

for all i and j . ¯ and define the Hence only two terms of (5.2) are not zero. Moreover, since same polarization at each Fi one of these terms can be modified using ¯

Res (IFεi ) = Res (IFεi ). Hence these computations transform (5.2) into ¯ ε )= Res (IFεi ). Res− (IM 0

(5.3)

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Let us now take the limit of both sides of (5.3) as ε → 0. By property (3) of the residue map, and by equations (3.16) and (4.8), we have ¯ ε lim Res− (IM ) = c κ0 (ηeω ), 0 ε→0+

for some constant

M0

c .

M0

Hence the limit of (5.3) gives ' ω iµ (Fi ) e κ0 (ηe ) = c Res i

ι∗Fi (η eω ) Fi

*

e(ν(Fi ))

for some constant c. To finish the proof of Theorem A, remember that Fi are the old connected components of the fixed point set MT , so that Fi ⊂ M T and µ(Fi ) = µ (Fi ). In particular, ι∗Fi (η eω ) is the same as the restriction of ηeω ∈ HT∗ (M) to Fi . Moreover, if for a connected component F of M T its moment map image µ(F ) is not inside , then the cone at F polarized with respect to does not contain the origin, and by property (1) of the residue the term which corresponds to F in the formula (1.1) is zero.

References [A]

M. F. Atiyah, Convexity and commuting Hamiltonians, Bull. London Math. Soc., 14 (1982), 1–15. [AB] M. F. Atiyah and R. Bott, The moment map and equivariant cohomology, Topology, 23-1 (1984), 1–28. [BV] N. Berline and M. Vergne, Classes caractéristiques équivariantes: Formule de localisation en cohomologie équivariante, C. R. Acad. Sci. Paris Sér. I Math., 295-9 (1982), 539–541. [BT] R. Bott and L. Tu, Differential Forms in Algebraic Topology, Springer-Verlag, New York, 1982. [BGL] D. Burns, V. Guillemin, and E. Lerman, Kähler cuts, arXiv:math.DG/ 0212062. [Go] R. F. Goldin, An effective algorithm for the cohomology ring of symplectic reductions, Geom. Functional Anal., 12 (2002) 567–583 [GK] V. Guillemin and J. Kalkman, The Jeffrey–Kirwan localization theorem and residue operations in equivariant cohomology, J. Reine Angew. Math., 470 (1996), 123–142. [GS] V. Guillemin and S. Sternberg, Convexity properties of the moment mapping I, Invent. Math., 67 (1982), 491–513. [JK1] L. C. Jeffrey and F. C. Kirwan, Localization for nonabelian group actions, Topology, 34-2 (1995), 291–327. [JK2] L. C. Jeffrey and F. C. Kirwan, Localization and the quantization conjecture, Topology, 36-3 (1997), 647–693. [K] F. Kirwan, Cohomology of Quotients in Symplectic and Algebraic Geometry, Princeton University Press, Princeton, NJ, 1984. [Le] E. Lerman, Symplectic cuts, Math. Res. Lett., 2-3 (1995), 247–258. [LMTW] E. Lerman, E. Meinrenken, S. Tolman, and C. Woodward, Nonabelian convexity by symplectic cuts, Topology, 37-2 (1998), 245–259. [Me] E. Meinrenken, Symplectic surgery and the Spin-c Dirac operator, Adv. Math., 134 (1998), 240–277

Refinements of the Morse stratification of the normsquare of the moment map∗ Frances Kirwan Mathematical Institute Oxford University Oxford OX1 3LB UK [email protected] This paper is dedicated to Alan Weinstein with many thanks and best wishes on the occasion of his 60th birthday. Abstract. Let X be any nonsingular complex projective variety on which a complex reductive group G acts linearly, and let Xss and Xs be the sets of semistable and stable points of X in the sense of Mumford’s geometric invariant theory GIT [17]. Then X has a G-equivariantly perfect stratification by locally closed nonsingular G-invariant subvarieties with Xss as an open stratum, which can be obtained as the Morse stratification of the normsquare of a moment map for the action of a maximal compact subgroup K of G [9]. In this paper this stratification is refined to obtain stratifications of X by locally closed nonsingular G-invariant subvarieties with X s as an open stratum. The strata can be defined inductively in terms of the sets of stable points of closed nonsingular subvarieties of X acted on by reductive subgroups of G and their projectivized normal bundles. When G is abelian, another way to obtain a refined stratification is by perturbing the moment map; the refinement is then itself equivariantly perfect, and its strata can be described in terms of the sets of stable points of linear actions of reductive subgroups of G for which semistability and stability coincide. This is useful even when G is nonabelian, since important questions about the cohomology of the GIT quotient (or Marsden–Weinstein reduction) X//G can be reduced to questions about the quotient of X by a maximal torus of G.

Let X be any nonsingular complex projective variety with a linear action of a complex reductive group G, and let Xss and X s be the sets of semistable and stable points of X in the sense of Mumford’s geometric invariant theory [17]. We can choose a maximal compact subgroup K of G and an inner product on the Lie algebra k of K which is invariant under the adjoint action. Then X has a G-equivariantly perfect stratification {Sβ : β ∈ B} by locally closed nonsingular G-invariant subvarieties with X ss as an ∗ The author is a member of VBAC (Vector Bundles on Algebraic Curves), which is par-

tially supported by EAGER (EC FP5 contract HPRN-CT-2000-00099), and acknowledges with gratitude the hospitality of the University of Melbourne and the Australian National University during the writing of part of this paper.

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open stratum, which can be obtained as the Morse stratification for the normsquare of a moment map µ : X → k∗ for the action of K on X [9]. In this note the Morse stratification {Sβ : β ∈ B} is refined to obtain stratifications of X by locally closed nonsingular G-invariant subvarieties with X s as an open stratum. The strata can be defined inductively in terms of the sets of stable points of closed nonsingular subvarieties of X acted on by reductive subgroups of G, and their projectivized normal bundles. These refinements of the Morse stratification are not in general equivariantly perfect; that is, the associated equivariant Morse inequalities are not necessarily equalities. However, when G is abelian, we can modify the moment map (or equivalently modify the linearisation of the action) by the addition of any constant since the adjoint action is trivial. Perturbation of the moment map by adding a small constant then provides an equivariantly perfect refinement of the stratification {Sβ : β ∈ B}, and a generic perturbation gives us a refined stratification whose strata can be described inductively in terms of the sets of stable points of linear actions of reductive subgroups of G for which stability and semistability coincide. This is useful even when G is not abelian, since important questions about the cohomology of the Marsden– Weinstein reduction µ−1 (0)/K (or equivalently the geometric invariant theoretic quotient X//G) can be reduced to questions about the quotient of X by a maximal torus of G. The same constructions work when X is a compact Kähler manifold with a Hamiltonian action of K. Even when X is symplectic but not Kähler, refinements of the Morse stratification for µ2 can be obtained by choosing a suitable almost complex structure and Riemannian metric. The moduli spaces M(n, d) of holomorphic bundles of rank n and degree d over a Riemann surface of genus g ≥ 2 can be constructed as quotients of infinitedimensional spaces of connections in a way that is analogous to the construction of quotients in geometric invariant theory; the role of the moment map is played by curvature and the role of the normsquare of the moment map is played by the Yang– Mills functional. In [13] refinements of the Morse stratification of the Yang–Mills functional are studied using the ideas of this paper. The motivation for this study was the search for a complete set of relations among the standard generators for the cohomology of these moduli spaces M(n, d) when n and d are coprime and n > 2 [4]. The layout of this paper is as follows. Section 1 reviews some background material and Section 2 uses the partial desingularisation construction of [10] to define a stratification {γ : γ ∈ } of Xss with X s as an open stratum. Section 3 gives an inductive description of the strata γ in X ss in terms of the stable and semistable points of linear actions of reductive subgroups and subquotients of G on nonsingular subvarieties of X and their projectivized normal bundles. Section 4 refines the stratification {γ : γ ∈ } to obtain strata which are described inductively purely in terms of the stable points (not the semistable points) of the linear actions appearing in Section 3, and in Section 5 this stratification is used to refine the Morse stratification {Sβ : β ∈ B} of X. In Section 6 an alternative refinement of this stratification is obtained when G is abelian by perturbing the moment map; in this case the inner product on the Lie algebra of K can also be perturbed to give a refined stratification.

Morse stratification of the normsquare of the moment map

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Finally Section 7 discusses applications to the study of the cohomology ring of the Marsden–Weinstein reduction µ−1 (0)/K (or equivalently the geometric invariant theoretic quotient X//G), and in particular the relationship between this cohomology ring and the corresponding cohomology ring when G is replaced by a maximal torus.

1 Background In this section we shall review briefly the material we need from [9] (see also [6, 17, 18]). Let X be a connected nonsingular projective variety embedded in projective space Pn and let G be a complex reductive group acting linearly on X via a homomorphism ρ : G → GL(n + 1; C). Then G is the complexification of a maximal compact subgroup K, and by rechoosing the coordinates on Pn if necessary, we can assume that K acts unitarily on Pn via ρ : K → U (n + 1). The geometric invariant theoretic quotient X//G is the projective variety whose homogeneous coordinate ring is the G-invariant part of the homogeneous coordinate ring of X. A point x of X is called semistable if there exists an invariant homogeneous polynomial f which does not vanish on x, and x is called stable if in addition the orbit Gx is a closed subset of the set of semistable points X ss and has dimension dim G. There is a rational map from X to X//G which restricts to a G-invariant surjective morphism φ : Xss → X//G from the open subset Xss of X, and every fibre of φ which meets the set X s consisting of the points of X which are stable for the action of G is a single G-orbit in Xss . The image of Xs is an open subset of X//G which can thus be identified via φ with the quotient X s /G. We shall assume that X s = ∅ (but see Remark 2.1). X has a Kähler structure given by the restriction of the Fubini–Study metric on Pn , and the Kähler form ω is a K-invariant symplectic form in X. There is a moment map µ : X → k∗ , where k is the Lie algebra of K, defined by µ(x) = ρ ∗ ((2π ix ∗ 2 )−1 x ∗ x¯ ∗t ) for x ∈ X ⊆ Pn represented by x ∗ ∈ Cn+1 \{0}, when the Lie algebra of U (n + 1) and its dual are both identified with the space of skew-Hermitian (n + 1) × (n + 1) matrices in the standard way. Then µ−1 (0) is a subset of Xss , and the inclusion induces a homeomorphism from the Marsden–Weinstein reduction (or symplectic quotient) µ−1 (0)/K to the geometric invariant theoretic quotient X//G. In fact, X ss is the set of points x in X such that µ−1 (0) meets the closure of the G-orbit of x, and X s is the set of points x in X such that µ−1 (0) meets the G-orbit of x at a point which is regular for µ. In the good case when Xss = Xs then X//G = X ss /G and its rational cohomology is isomorphic to the equivariant cohomology of X ss . If we fix an invariant inner product on the Lie algebra k, then we can consider the function µ2 as a Morse function on X. It is not in general a Morse function in the classical sense, or even a Morse–Bott function, since the connected components of

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its set of critical points may not be submanifolds of X, but nonetheless it induces a Morse stratification {Sβ : β ∈ B} of X such that the stratum to which x ∈ X belongs is determined by the limit set of its path of steepest descent for µ2 with respect to the Fubini–Study metric. This stratification can also be defined purely algebraically and has the following properties [9]. Proposition 1.1. (i) Each stratum Sβ is a G-invariant locally closed nonsingular subvariety of X. (ii) The unique open stratum S0 is the set X ss of semistable points of X. (iii) The stratification is equivariantly perfect over the rationals, so that i−λ(β) dim HG (Sβ ), dim HGi (X) = dim HGi (X ss ) + β=0

where λ(β) is the real codimension of Sβ in X. (iv) If β = 0, then there is a proper nonsingular subvariety Zβ of X acted on by a reductive subgroup Stab β of G such that ∗ (Zβss ), HG∗ (Sβ ) ∼ = HStab(β)

where Zβss is the set of semistable points of Zβ with respect to an appropriate linearisation of the action of Stab(β). Remark 1.2. (i) All cohomology in this paper has rational coefficients. (ii) We shall assume that the invariant inner product chosen on k is rational, and we shall use it to identify k∗ with k throughout. (iii) Note that G-equivariant cohomology is the same as K-equivariant cohomology, since G retracts onto its maximal compact subgroup K. If we choose a positive Weyl chamber t+ in the Lie algebra t of a maximal torus T of K, then we can identify the indexing set B with a finite subset of t+ (or equivalently with the set of adjoint orbits of the points in this finite subset of t+ , since each adjoint orbit meets t+ at exactly one point). More precisely, let α0 , . . . , αn be the weights of the representation of T on Cn+1 and use the restriction to t of the fixed invariant inner product on k to identify t∗ with t. Then β ∈ t+ belongs to B if and only if β is the closest point to 0 of the convex hull in t of some nonempty subset of {α0 , . . . , αn }. Moreover, Stab(β) is the stabiliser of β under the adjoint action of G, and Zβ is the intersection of X with the linear subspace {[x0 : · · · : xn ] ∈ Pn : xi = 0 if αi .β = β2 } of Pn . Equivalently, Zβ is the union of those connected components of the fixed point set of the subtorus Tβ of T generated by β on which the constant value taken by the real-valued function x → µ(x).β is β2 . If we use the fixed inner product to identify k with its dual, then the image µ(Zβ ) of Zβ is contained in the Lie algebra of


331

the maximal compact subgroup StabK (β) = K ∩ Stab(β) of Stab(β). Since moment maps are only unique up to the addition of a central constant, we can take µ − β as our moment map for the action of StabK (β) on Zβ . This corresponds to a modification of the linearisation of the action of Stab(β) on Zβ whose restriction to the complexification Tβc of Tβ is trivial, and we define Zβss to be the set of semistable points of Zβ with respect to this modified linear action. Equivalently, Zβss is the stratum labelled by 0 (the minimum stratum) for the Morse stratification of the function µ − β2 on Zβ . Then A Sβ = GY¯β \ GY¯γ = GYβss , (1.1) γ >β

where Y¯β = {x ∈ X : xi = 0 if αi .β < β2 } and Yβ = {x ∈ Y¯β : xi = 0 for some i such that αi .β = β2 }, while

Yβss = pβ−1 (Zβss ),

(1.2)

where pβ : Yβ → Zβ is the obvious projection given by pβ (x) = lim exp(−itβ)x. t→∞

(1.3)

Remark 1.3. In [9] Zβss is defined as above to be the set of semistable points of Zβ with respect to the action of Stab(β) with the linearisation modified in a way which corresponds to replacing the moment map µ by (a positive integer multiple of) µ − β. However, we can, if we wish, regard µ − β as a moment map for the action of StabK (β)/Tβ on Zβ , and then Zβss is the set of semistable points for the induced linear action of its complexification Stab(β)/Tβc . The advantage of this description is that the analogous definition of Zβs is a useful one, whereas Zβ has no points that are stable with respect to the action of Stab(β) when β = 0. Therefore, we shall define Zβs to be the set of stable points for the action of Stab(β)/Tβc on Zβ , linearized so that the corresponding moment map is a positive integer multiple of µ − β. Equivalently, Zβss and Zβs are the sets of semistable (respectively, stable) points of Zβ under the action of the subgroup of Stab(β) whose Lie algebra is the complexification of the orthogonal complement to β in the Lie algebra of StabK (β). In fact, if B is the Borel subgroup of G associated to the choice of positive Weyl chamber t+ and if Pβ is the parabolic subgroup B Stab(β), then Yβ and Yβss are Pβ -invariant and we have Sβ ∼ (1.4) = G ×Pβ Yβss . Moreover, Yβ is a nonsingular subvariety of X and pβ : Yβ → Zβ is a locally trivial fibration whose fibre is isomorphic to Cmβ for some mβ ≥ 0.

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Now an element g of G lies in the parabolic subgroup Pβ if and only if exp(−itβ)g exp(itβ) tends to a limit in G as t → ∞, and this limit defines a surjection qβ : Pβ → Stab(β). Since the surjections pβ : Yβss → Zβss and qβ : Pβ → Stab(β) are retractions satisfying pβ (gx) = qβ (g)pβ (x) (1.5) for all g ∈ Pβ and x ∈ Yβss , this gives us the isomorphism ∗ (Zβss ) HG∗ (Sβ ) ∼ = HStab(β)

of Proposition 1.1(iv). Moreover, since G = KB and B ⊆ Pβ we have GY¯β = K Y¯β , which is compact, and hence A S¯β ⊆ GY¯β ⊆ Sβ ∪ Sγ . (1.6) γ >β

Note that x = [x0 , . . . , xn ] ∈ X is semistable (respectively stable) for the action of the complex torus T c if and only if 0 belongs to the convex hull in t of the set of weights {αj : xj = 0} (respectively to the interior of this convex hull), and that x is semistable (respectively stable) for the action of G if and only if every element gx of its G-orbit is semistable (respectively stable) for the action of T c . In particular this tells us that S0 = Xss . It also tells us that if β ∈ B and y ∈ Y¯β \Y ss , then there is a subset S of {αj : αj .β ≥ β

β2 } such that where

β

y ∈ Stab(β)Yβ ,

is the closest point to 0 of the convex hull of S and

(1.7) β

= β.

Remark 1.4. Of course, the definitions of the subvarieties Zβ , Zβss and so on in this section depend on the action of G on X ⊆ Pn and its linearisation via the representation ρ : G → GL(n + 1; C). When it is necessary to make these explicit in the notation we shall write Zβ (X, ρ), Zβss (X, ρ) and so on, but we shall omit X if X = Pn , so that, for example, Zβ (X, ρ) = X ∩ Zβ (ρ). Remark 1.5. In the special case when every semistable point is stable, the quotient variety X//G is topologically the ordinary quotient Xss /G, where G acts with only finite stabilisers on Xss , which means that its Betti numbers dim H i (X//G) are the same as the equivariant Betti numbers dim HGi (X ss ) of Xss . These can be calculated inductively using Proposition 1.1 together with the fact that the equivariant cohomology of a nonsingular complex projective variety is isomorphic as a vector space to the tensor product of its ordinary cohomology and the equivariant cohomology of a point. Remark 1.6. If X is any compact symplectic manifold with a Hamiltonian action of a compact Lie group K and a moment map µ : X → k∗ , then the Morse stratification of µ2 has essentially the properties described here, with G replaced by K and Pβ replaced by K ∩ Stab(β) [9].


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2 Stratifying the set of semistable points Suppose now that X has some stable points but also has semistable points that are not stable. In [10, 11] it is described how one can blow X up along a sequence of nonsingular G-invariant subvarieties to obtain a G-invariant morphism X˜ → X, where X˜ is a complex projective variety acted on linearly by G such that X˜ ss = X˜ s . ˜ The induced birational morphism X//G → X//G of the geometric invariant theoretic ˜ quotients is then a partial desingularisation of X//G in the sense that X//G has only orbifold singularities (it is locally isomorphic to the quotient of a nonsingular variety by a finite group action) whereas the singularities of X//G are in general much worse. In this section we shall review the construction of the partial desingularisation ˜ X//G and use it firstly to stratify Xss and subsequently (in Section 5) to refine the stratification {Sβ : β ∈ B} of X described in Section 1. The set X˜ ss can be obtained from X ss as follows. There exist semistable points of X that are not stable if and only if there exists a nontrivial connected reductive subgroup of G fixing a semistable point. Let r > 0 be the maximal dimension of a reductive subgroup of G fixing a point of X ss and R(r) a set of representatives of conjugacy classes of all connected reductive subgroups R of dimension r in G such that ZRss = {x ∈ Xss : R fixes x} is nonempty. Then

A

GZRss

R∈R(r)

is a disjoint union of nonsingular closed subvarieties , of X ss . The action of G on ss ss X lifts to an action on the blowup X(1) of X along R∈R(r) GZRss which can be ss in X linearized so that the complement of X(1) (1) is the proper transform of the subset φ −1 (φ(GZRss )) of Xss , where φ : X ss → X//G is the quotient map (see [10, 7.17]). ss is fixed by a reductive subgroup of G of dimension at Moreover, no point of X(1) ss least r, and a point in X(1) is fixed by a reductive subgroup R of dimension less than r in G if and only if it belongs to the proper transform of the subvariety ZRss of X ss . ss to obtain X ss such that no reductive We can now apply the same procedure to X(1) (2) ss . If we repeat this process subgroup of G of dimension at least r −1 fixes a point of X(2) ss = X ss , X ss , X ss , . . . , X ss such that no reductive enough times, we obtain X(0) (1) (2) (r) ss , and we set X ˜ ss = Xss . subgroup of G of positive dimension fixes a point of X(r) (r) Equivalently, we can construct a sequence ss ss ss X(R = X ss , X(R , . . . , X(R = X˜ ss , τ) 0) 1)

where R1 , . . . , Rτ are connected reductive subgroups of G with r = dim R1 ≥ dim R2 ≥ · · · dim Rτ ≥ 1, ss along its closed nonsingular and if 1 ≤ l ≤ τ , then X(Rl ) is the blow up of X(R l−1 ) ss ss subvariety GZRl ∼ = G ×Nl ZRl , where Nl is the normaliser of Rl in G. Similarly,

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˜ X//G = X˜ ss /G can be obtained from X//G by blowing up along the proper transforms of the images ZR //N in X//G of the subvarieties GZRss of Xss in decreasing order of dim R. If 1 ≤ l ≤ τ , then there is a G-equivariant stratification {Sβ,l : β ∈ Bl } of X(Rl ) by nonsingular G-invariant locally closed subvarieties such that one of the ss of X . This stratification strata, indexed by 0 ∈ Bl , coincides with the open subset XR Rl l is constructed exactly as the stratification {Sβ : β ∈ B} of X was constructed in the last section; note that X(Rl ) is in general only quasi-projective rather than projective, but it is shown in [10] that the construction of the stratification still works for X(Rl ) and the properties given in Proposition 1.1 still hold. There is a partial ordering on Bl with 0 as its minimal element such that if β ∈ Bl , then the closure in X(Rl ) of the stratum Sβ,l satisfies Sβ,l ⊆

A

Sγ ,l .

γ ∈Bl ,γ ≥β

If β ∈ Bl and β = 0, then the stratum Sβ,l retracts G-equivariantly onto its (tranverse) ss intersection with the exceptional divisor El for the blowup X(Rl ) → X(R . This l−1 ) ss ˆ exceptional divisor is isomorphic to the projective bundle P(Nl ) over GZ , where Rl

ss Zˆ Rssl is the proper transform of ZRssl in X(R and Nl is the normal bundle to GZˆ Rssl l−1 ) ss in XRl−1 . The stratification {Sβ,l : β ∈ Bl } is determined by the action of Rl on the fibres of Nl over ZRssl (see [10, Section 7]). The composition ss ss ss → X(R → · · · X(R → X ss X˜ ss = X(R τ) τ −1 ) 1)

is an isomorphism over the set X s of stable points of X, and the complement of X s in X˜ ss is just the union of the proper transforms in X˜ ss of the exceptional divisors ss E1 , . . . , Ek for the blowups XRl → X(R for l = 1, . . . , τ . l−1 ) ss We can now stratify X as follows. We take as the highest stratum the nonsingular closed subvariety GZRss1 whose complement in Xss can be naturally identified with the complement X(R1 ) \E1 of the exceptional divisor E1 in X(R1 ) . Recall that GZRss1 ∼ = G ×N1 ZRss1 , where N1 is the normaliser of R1 in G, and ZRss1 is equal to the set of semistable points for the action of N1 , or equivalently for the induced action of N1 /R1 , on ZR1 , which is a union of connected components of the fixed point set of R1 in X (see [10, Section 5]). Since R1 has maximal dimension among those reductive subgroups of G with fixed points in Xss , we have ZRss1 = ZRs 1 , where ZRs l is the set of stable points for the action of Nl /Rl on ZRl for 1 ≤ l ≤ τ . Next, we take as strata the nonsingular locally closed subvarieties


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{Sβ,1 \E1 : β ∈ B1 , β = 0} ss \E of X(R1 ) \E1 = X ss \GZRss1 , whose complement in X(R1 ) \E1 is X(R 1 = 1) ss ss ss ss ss \E X(R1 ) \E1 , where E1 = X(R1 ) ∩ E1 , and then we take the intersection of X(R 1 1) with GZRss2 . This intersection is GZRs 2 , where ZRs 2 is the set of stable points for the ss \E can be naturally identified action of N2 /R2 on ZR2 , and its complement in X(R 1 1) with the complement in X(R2 ) of the union of E2 and the proper transform Eˆ 1 of E1 . Our next strata are the nonsingular locally closed subvarieties

{Sβ,2 \(E2 ∪ Eˆ 1 ) : β ∈ B2 , β = 0} ss \(E ∪ E ˆ 1 ), of X(R2 ) \(E2 ∪ Eˆ 1 ), whose complement in X(R2 ) \(E2 ∪ Eˆ 1 ) is X(R 2 2) s and the stratum after these is GZR3 . Repeating this process gives us strata that are all nonsingular locally closed G-invariant subvarieties of X ss indexed by the disjoint union {R1 } ∪ {R1 } × (B1 \{0}) ∪ · · · ∪ {Rτ } ∪ {Rτ } × (Bτ \{0}),

and the complement in Xss of the union of these strata is just the open subset X s . We take Xs as our final stratum indexed by 0, so that the indexing set for our stratification of Xss is the disjoint union = {R1 } ∪ {R1 } × (B1 \{0}) ∪ · · · ∪ {Rτ } ∪ {Rτ } × (Bτ \{0}) ∪ {0}.

(2.1)

Moreover, the given partial orderings on B1 , . . . , Bτ together with the ordering in the expression (2.1) above for induce a partial ordering on , with R1 as the maximal element and 0 as the minimal element, such that the closure in Xss of the stratum γ indexed by γ ∈ satisfies A γ ⊆ δ . (2.2) δ∈,δ≥γ

Thus this process gives us a stratification {γ : γ ∈ }

(2.3)

of Xss such that the stratum indexed by the minimal element 0 of coincides with the open subset X s of X ss . Remark 2.1. We have been assuming that X s = ∅, but this procedure gives us a stratification of X ss even when X s is empty. The only difference when X s is empty is that the procedure terminates at some stage l when ss X(R = GZˆ Rssl ∼ = G ×Nl Zˆ Rssl l−1 )

and gives us a stratification indexed by = {R1 } ∪ {R1 } × (B1 \{0}) ∪ · · · ∪ {Rl−1 } ∪ {Rl−1 } × (Bl−1 \{0}) ∪ {Rl } such that the stratum indexed by the minimal element Rl of is the open subset GZRs l of X ss . Note also that ZRs l is nonempty, since otherwise

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ZRssl = Nl ZRss for some R containing Rl with dim R > dim Rl , and then GZRss = GZRss = X ss , so the procedure would have terminated at an earlier stage.

3 Inductive description of the strata γ in Xss The last section described a stratification {γ : γ ∈ } of X ss such that the stratum indexed by the minimal element 0 of coincides with the open subset X s of X ss . In this section we shall study the strata γ in more detail. Note that the strata γ with γ = 0 fall into two classes. Either γ = Rl for some l ∈ {1, . . . , τ }, in which case the stratum γ is GZRs l , or else γ = (Rl , β), where β ∈ Bl \{0} for some l ∈ {1, . . . , τ } and the stratum γ is Sβ,l \(El ∪ Eˆ l−1 ∪ · · · ∪ Eˆ 1 ). In the latter case, we know from (1.4) that ss ∼ ss Sβ,l = GYβ,l , = G ×Pβ,l Yβ,l

(3.1)

ss fibres over Z ss via p : Y ss → Z ss with fibre Cmβ,l for some m where Yβ,l β β,l > β,l β,l β,l 0, and ss ss Sβ,l ∩ El = G(Yβ,l ∩ El ) ∼ ∩ El ), (3.2) = G ×Pβ,l (Yβ,l ss ∩ E fibres over Z ss with fibre Cmβ,l −1 (see [10, Lemmas 7.6 and 7.11]). where Yβ,l l β,l Thus ss Sβ,l \El ∼ \El ), (3.3) = G ×Pβ,l (Yβ,l ss \E fibres over Z ss with fibre Cmβ,l −1 × (C\{0}). Let where Yβ,l l β,l

πl : El ∼ = P(Nl ) → GZˆ Rssl denote the projection. [10, Lemma 7.9] tells us that if x ∈ Zˆ Rssl , then the intersection of Sβ,l with the fibre πl−1 (x) = P(Nl,x ) of πl at x is the union of those strata indexed by points in the adjoint orbit Ad(G)β in the stratification of P(Nl,x ) induced by the representation ρl of Rl on the normal Nl,x to GZˆ Rssl at x. Note that we can assume that Rl ∩ K is a maximal compact subgroup of Rl and that Rl ∩ T is a maximal torus for Rl ∩ K, and then Ad(G)β meets a positive Weyl chamber for Rl in Lie(Rl ∩ T ) in a finite number of points


β = β1 = Ad(w1 )β,

β2 = Ad(w2 )β,

...,

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βrβ,l = Ad(wrβ,l )β,

where w1 = 1, w2 , . . . , wrβ,l ∈ G represent elements of the Weyl group of G. ss and π (y) = gx, where g ∈ G and x ∈ Z ˆ ss , then x is fixed by Now if y ∈ Zβ,l l Rl −1 −1 Ad(g )β and so Ad(g )β lies in the Lie algebra of Rl . Since Rl ∩ T is a maximal compact torus of Rl , there exists r ∈ Rl such that Ad(rg −1 )β ∈ Lie(Rl ∩ T ). Then Ad(rg −1 )β = Ad(wj )β for some j ∈ {1, . . . , rβ,l }, and hence wj−1 rg −1 ∈ Stab(β),

so g ∈ Stab(β)wj−1 Rl . Conversely if g = hwj−1 r, where h ∈ Stab(β) and r ∈ Rl , ss if and only if h−1 y lies in Z ss , where π (h−1 y) = w −1 rx ∈ w −1 Z ˆ ss . then y ∈ Zβ,l l β,l Rl j j Thus

A ss ss = Stab(β) Zβ,l ∩ wj−1 πl−1 (Zˆ Rssl ) Zβ,l 1≤j ≤rβ,l

=

A

1≤j ≤rβ,l

−1 ˆ ss ss Stab(β)wj−1 ZAd(w ∩ π ( Z ) . Rl l j )β,l

ss ∩ w −1 π −1 (Z ˆ ss )) meets Stab(β)(Z ss ∩ w −1 π −1 (Zˆ ss )), then Also, if Stab(β)(Zβ,l Rl β,l Rl j l i l Stab(β)wj−1 Zˆ Rssl meets wi−1 Zˆ Rssl , and since GZˆ Rssl ∼ = G ×Nl Zˆ Rssl , this means that there is some h ∈ Stab(β) and n ∈ Nl such that wi h = nwj , so that βi = Ad(wi )β ∈ Ad(Nl )βj . Conversely, if βi ∈ Ad(Nl )βj then wi h = nwj for some h ∈ Stab(β) and n ∈ Nl , and so ss ss Stab(β)(Zβ,l ∩ wj−1 πl−1 (Zˆ Rssl )) = Stab(β)(Zβ,l ∩ h−1 wi−1 nπl−1 (Zˆ Rssl )) ss = Stab(β)(Zβ,l ∩ wi−1 πl−1 (Zˆ Rssl )). ss is a disjoint union Thus Zβ,l ss Zβ,l =

B

ss Stab(β) Zβ,l ∩ wj−1 πl−1 (Zˆ Rssl ) ,

1≤j ≤sβ,l

where Ad(w1 )β = β, . . . , Ad(wsβ,l )β form a set of representatives for the Ad(Nl ) ss and S orbits in Ad(G)β, and Yβ,l β,l can be expressed similarly as disjoint unions. In fact, since by (1.5) the fibration ss ss pβ : Yβ,l → Zβ,l ss , where q : P → satisfies pβ (gy) = qβ (g)pβ (y) for all g ∈ Pβ and y ∈ Yβ,l β β Stab(β) is the projection, we have

B ss ss Yβ,l = Pβ pβ−1 Zβ,l ∩ wj−1 πl−1 (Zˆ Rssl ) 1≤j ≤sβ,l

and

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B

Sβ,l =

ss Gpβ−1 Zβ,l ∩ wj−1 πl−1 (Zˆ Rssl ) .

1≤j ≤sβ,l

This means that we could, if we wished, replace the indexing set Bl \{0}, whose elements correspond to the G-adjoint orbits Ad(G)β of elements of the indexing set for the stratification of P(Nl,x ) induced by the representation ρl , by the set of their Nl -adjoint orbits Ad(Nl )β. Then we would still have (3.1)–(3.3), but now ss ss ss = Stab(β)(Zβ,l ∩ πl−1 (Zˆ Rssl )) ∼ ∩ πl−1 (Zˆ Rssl )) (3.4) Zβ,l = Stab(β) ×Nl ∩Stab(β) (Zβ,l

and

ss ∼ ss ∩ wj−1 πl−1 (Zˆ Rssl )), Yβ,l = Pβ ×Qβ pβ−1 (Zβ,l

where

(3.5)

Qβ = qβ−1 (Nl ∩ Stab(β))

is a subgroup of Pβ , and hence

ss ∼ ss Sβ,l ∼ ∩ wj−1 πl−1 (Zˆ Rssl ) . = G ×Pβ Yβ,l = G ×Qβ pβ−1 Zβ,l

(3.6)

Furthermore, πl now restricts to a fibration ss ∩ πl−1 (Zˆ Rssl )) → Zˆ Rssl πl : Zβ,l

(3.7)

whose fibre at x ∈ Zˆ Rssl is Zβss (ρl ) defined as in Remark 1.4, where ρl is the representation of Rl on the normal Nl,x to GZˆ ss at x. Rl

ss of the exceptional If 1 ≤ j ≤ l − 1, then the proper transform Eˆ j in X(R l) ss meets the exceptional divisor E ∼ P(N ) transversely, divisor Ej in X(R and their = l l ) j intersection is the restriction P(Nl |Eˆ j ∩GZˆ R ) l

ss of the projective bundle P(Nl ) over GZˆ Rssl to the intersection in X(R of GZˆ Rssl with l−1 ) ss the proper transform of Ej in X(Rl−1 ) (which by abuse of notation we shall also denote by Eˆ j ). Moreover, the complement in GZˆ ss of its intersection with the exceptional

divisors Eˆ 1 , . . . , Eˆ l−1 is GZRs l . Thus

Rl

\E \E γ = GYβ,l ∼ = G ×Pβ Yβ,l ,

where

(3.8)

\E

ss \(El ∪ Eˆ l−1 ∪ · · · ∪ Eˆ 1 ) Yβ,l = Yβ,l

ss ∩ π −1 (Z s )) with fibre Cmβ,l −1 × (C\{0}), and fibres over Stab(β) ×Nl ∩Stab(β) (Zβ,l Rl l

ss ∩ π −1 (Z s ) fibres over Z s ss Zβ,l Rl l (Rl ) with fibre Zβ (ρl ). In addition, if we set

\E \E ss Yβ = Yβ,l ∩ pβ−1 Zβ,l ∩ πl−1 (Zˆ Rssl ) ,


339

we have from (3.5) and (3.6) that

and hence

\E \E Yβ,l ∼ = Pβ ×Qβ Yβ

(3.9)

\E γ ∼ = G ×Qβ Yβ ,

(3.10)

\E

where Qβ = qβ−1 (Nl ∩ Stab(β)) and pβ : Yβ with fibre Cmβ,l −1 × (C\{0}).

ss ∩ π −1 (Z ˆ ss ) is a fibration → Zβ,l Rl l

Remark 3.1. The moduli space M(n, d) of semistable holomorphic bundles of rank n and degree d over a fixed Riemann surface of genus g ≥ 2 can be constructed as a quotient of an infinite-dimensional affine space of connections C by a complexified gauge group Gc , in an infinite-dimensional version of the construction of quotients in geometric invariant theory, or, equivalently, as an infinite-dimensional symplectic reduction with curvature as a moment map. When n and d are coprime, semistability coincides with stability and M(n, d) is the topological quotient of the semistable subset C ss of C by the action of Gc . The role of the normsquare of the moment map is played by the Yang–Mills functional, which was studied by Atiyah and Bott in their fundamental paper [1]. Atiyah and Bott studied the stratification of C defined using the Harder–Narasimhan type of holomorphic bundle, which they expected to be the Morse stratification of the Yang–Mills functional (this was later shown to be the case [2]). The methods of this paper can be used to provide a stratification {γ : γ ∈ } of C ss with C s as the unique open stratum. This stratification of C ss and induced refinements of the Yang–Mills stratification of C are studied in detail in [13], where they are related to natural refinements of the notion of the Harder–Narasimhan type of a holomorphic bundle.

4 A refined stratification of Xss We can now iterate the construction of the stratification (2.3) described in Section 2 and use induction on the dimension of G to define a stratification ˜ ˜ γ˜ : γ˜ ∈ } {

(4.1)

of Xss by G-equivariant nonsingular subvarieties which refines the stratification (2.3). When the dimension of G is zero so that X s = X ss = X, then ˜ = and the stratification has one stratum which is X itself. When dim G > 0, we shall refine the stratification {γ : γ ∈ } defined in (2.3) as follows. If γ ∈ \{0, R1 , . . . , Rτ } then γ = (Rl , β), where β ∈ Bl \{0} for some l ∈ {1, . . . , τ }, and by (3.8) we have \E \E γ = GYβ,l ∼ = G ×Pβ Yβ,l , \E

ss ∩ π −1 (Z s )) with fibre Cmβ,l −1 × where Yβ,l fibres over Stab(β) ×Nl ∩Stab(β) (Zβ,l Rl l

ss ∩ π −1 (Z s ) fibres over Z s ss (C \ {0}), and Zβ,l Rl l (Rl ) with fibre Zβ (ρl ). We have a linear

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action of Rl ∩ Stab(β)/Tβc on Zβ (ρl ) which corresponds (up to multiplication by a positive integer) to the moment map µ − β. Therefore, by induction on dim G, we can ˜ γ : β˜ ∈ ˜ γ } of Z ss (ρl ) by nonsingular assume that we have defined a stratification { β β˜ Rl ∩ Stab(β)-invariant subvarieties. In fact, since the stabiliser in G of any x ∈ ZRs has connected component Rl , we can assume that we have a stratification of Zβss (ρl ) by nonsingular Stab(x) ∩ Stab(β)-invariant subvarieties. Since Stab(x) ⊆ Nl and since the fibration ss πl : Zβ,l ∩ πl−1 (ZRs l ) → ZRs l is Nl ∩ Stab(β)-equivariant with fibre Zβss (ρl ), this gives us a stratification of

ss ∩ π −1 (Z s ) by nonsingular N ∩ Stab(β)-invariant subvarieties, and hence a Zβ,l l Rl l stratification of ss Stab(β) ×Nl ∩Stab(β) (Zβ,l ∩ πl−1 (ZRs l ))

by nonsingular Stab(β)-invariant subvarieties. We also have a fibration \E ss ss \(El ∪ Eˆ l−1 ∪ · · · ∪ Eˆ 1 ) → Stab(β) ×Nl ∩Stab(β) (Zβ,l ∩ πl−1 (ZRs l )) pβ : Yβ,l = Yβ,l

with fibre Cmβ,l −1 × (C\{0}), which satisfies pβ (gx) = qβ (g)pβ (x) for all g ∈ Pβ \E \E and x ∈ Yβ,l (see (1.5)). Thus we get an induced stratification of Yβ,l by Pβ -invariant subvarieties, and finally an induced stratification of \E γ ∼ = G ×Pβ Yβ,l

˜ for β˜ ∈ ˜ γ . In particular γ has an open by nonsingular G-invariant subvarieties β˜ stratum ˜γ γs = (4.2) 0 γ

corresponding to the open stratum Zβs (ρl ) of Zβss (ρl ) consisting of stable points for the action of Rl ∩ Stab(β)/Tβc . ˜ γ˜ : γ˜ ∈ } ˜ of Xss indexed by In this way, we obtain a stratification { ˜ = {γ˜ = (γ ) : γ ∈ {0, R1 , . . . , Rτ }} ∪ {γ˜ = (Rl , β) : 1 ≤ l ≤ τ and β ∈ Bl \{0}} ∪ {γ˜ = (Rl , β, γ1 , . . . , γt ) : t ≥ 1 and 1 ≤ l ≤ τ and β ∈ Bl \{0} (4.3) and (γ1 , . . . , γt ) ∈ ˜ (Rl ,β) \{0}}, ˜ γ˜ are given by where ˜ (Rl ,β) is defined inductively as above, and the strata ˜ (0) = X s . If 1 ≤ l ≤ τ and β ∈ Bl \{0}, then ˜ (Rl ) = GZRs l

and

˜ (Rl ,β) = s (Rl ,β) ,

while if γ˜ = (Rl , β, γ1 , . . . , γt ), then ˜ (Rl ,β) . ˜ γ˜ = (γ1 ,...,γt )


341

5 The refined Morse stratification In Section 2 a stratification {γ : γ ∈ } of the set X ss of semistable points of X was defined, and in Section 4 this stratification was refined to give a stratification ˜ γ˜ : γ˜ ∈ } ˜ of X ss . Via the inductive description of the strata Sβ of the Morse {

stratification of µ2 in terms of the semistable points of nonsingular subvarieties of X given in Proposition 1.1, we can use these stratifications of X ss to refine the Morse stratification. ˜ γ˜ : γ˜ ∈ } ˜ of X ss conFor simplicity we shall just discuss the stratification { structed in Section 4. The construction of this stratification can be applied for each β ∈ B to the action of Stab(β) on the nonsingular projective subvariety Zβ of X that appeared in Proposition 1.1(iv) (or more precisely to the action of the quotient Stab(β)/Tβc of Stab(β) by its complex subtorus Tβc which acts trivially on Zβ ) to give a stratification ˜ [β] : γ˜ ∈ ˜ [β] } { γ˜

of Zβss by nonsingular Stab(β)-invariant subvarieties, with Zβs as the stratum indexed by (0). Since Sβ = GYβss satisfies (1.4) and we have a retraction pβ : Yβss → Zβss satisfying (1.5), we can stratify Sβ as the disjoint union of strata [β]

[β]

˜ )∼ ˜ ) Gpβ−1 ( = G ×Pβ pβ−1 ( γ˜ γ˜

(5.1)

for γ ∈ ˜ [β] . This gives us a stratification ˜ {S˜β˜ : β˜ ∈ B} of X indexed by

B˜ = ˜ ∪

A

(5.2)

{β} × ˜ [β] ,

β∈B\{0}

˜ ˜ defined as in Section 4 if β˜ ∈ , ˜ and if β˜ = (β1 , . . . , βt ), where where S˜β˜ = β β1 ∈ B\{0} and (β2 , . . . , βt ) ∈ ˜ [β] , then ˜ [β1 ] S˜β˜ = Gpβ−1 ( (β2 ,...,βt ) ). 1 ˜ refines the original stratification {Sβ : β ∈ B} and This stratification {S˜β˜ : β˜ ∈ B} has the following properties. Proposition 5.1. (i) Each stratum S˜β˜ is a G-invariant locally closed nonsingular subvariety of X. (ii) The unique open stratum S˜(0) is the set X s of stable points of X. ˜ then the closure S˜ ˜ in X (iii) There is a partial ordering > on B˜ such that if β˜ ∈ B, β ˜ of the stratum Sβ˜ satisfies A S˜β˜ ⊆ S˜γ˜ . γ˜ ≥β˜

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˜ ˜ and (iv) B˜ has a subset ˜ such that γ˜ < β˜ for all γ˜ ∈ ˜ and β˜ ∈ B\ A S˜γ˜ = X ss . γ˜ ∈˜

(v) If β˜ ∈ B˜ and β˜ = (0), then the stratum S˜β˜ can be described inductively in terms of the sets of stable points of certain nonsingular linear sections Z of X and projectivized normal bundles of nonsingular subvarieties of X, acted on by reductive subgroups of G and their quotients. Remark 5.2. If X is a compact Kähler manifold which has a Hamiltonian action of a compact group K with moment map µ : X → k∗ , then the Morse stratification for µ2 can be refined just as in Proposition 5.1. Even when X is symplectic but not Kähler we can construct a similar refinement by choosing a suitable almost complex structure and Riemannian metric on X (see [10, 16]). Example 5.3. Consider the action of G = SL(2; C) and its maximal compact subgroup K = SU (2) on X = (P1 )n , with the moment map given by the center of gravity in R3 when P1 is identified suitably with the unit sphere in R3 and R3 is identified with the Lie algebra of SU (2). An element (x1 , . . . , xn ) of (P1 )n is semistable (respectively stable) for the action of G if and only if at most n/2 (respectively strictly fewer than n/2) of the points xj coincide anywhere on P1 . The Morse stratification for the normsquare of the moment map on X has strata S0 = X ss and S2j −n for n/2 < j ≤ n. If n/2 < j ≤ n, then the elements of S2j −n correspond to sequences of n points on P1 such that exactly j of these points coincide somewhere on P1 , and S2j −n retracts equivariantly onto the subset of X, where j points coincide somewhere on P1 and the remaining n−j points coincide somewhere else on P1 , which is a single G-orbit with stabilizer C∗ , for j < n, and with stabiliser a Borel subgroup of G when j = n (see [9, Section 16.1] for more details). If n is odd, then semistability coincides with stability and the refined stratification coincides with the Morse stratification of X. that n is even, so that semistability and stability do not coincide. The semistable elements of X which are fixed by nontrivial connected reductive subgroups of G are those represented by sequences (x1 , . . . , xn ) of points of P1 such that there exist distinct p and q in P1 with exactly half of the points x1 , . . . , xn equal to p and the rest equal to q. They form n!/2((n/2)!)2 Gorbits, and their stabilisers are all conjugate to the maximal torus Tc = C∗ of G. These stabilisers act with weights 2 and −2, each with multiplicity (n/2) − 1, on ˜ the normals to the orbits. We obtain the partial desingularization X//G by blowing up X//G at the points corresponding to these orbits, or equivalently by blowing up X ss along these orbits, removing from the blowup the unstable points (which form the proper transform of the set of (x1 , . . . , xn ) ∈ X ss such that exactly half of the points x1 , . . . , xn coincide somewhere on P1 ) and finally quotienting by G. The ˜ of X thus has as its strata the set S˜(0) = X s of refined stratification {S˜β˜ : β˜ ∈ B} stable points, the set S˜(T ) consisting of points represented by sequences (x1 , . . . , xn ) in P1 such that there exist distinct p and q in P1 with exactly half of x1 , . . . , xn


343

equal to p and the rest equal to q, the set S˜(T ,2) consisting of points represented by sequences (x1 , . . . , xn ) in P1 such that there exists p in P1 with exactly half of the points x1 , . . . , xn equal to p and the rest different from p and not all equal to each other, and finally the strata S2j −n (for n/2 < j ≤ n) of the Morse stratification. Example 5.4. A very similar example is given by the action of G = SL(2; C) on X = Pn identified with the space of unordered sequences of n points in P1 ; that is, with the projectivized symmetric product P(S n (C2 )) (see [9, Section 16.2] for more details). The diagonal subgroup T ∼ = S 1 of K = SU (2) acts with weights n 2 n, n − 2, n − 4, . . . , 2 − n, −n on S (C ) = Cn+1 . An element [a0 , . . . , an ] of Pn corresponds to the n roots in P1 of the polynomial in one variable t with coefficients a0 , . . . , an ; it is semistable (respectively stable) for the action of G if and only if at most n/2 (respectively strictly fewer than n/2) of these roots coincide anywhere on P1 , and the Morse stratification for the normsquare of the moment map on X is essentially the same as in Example 5.3 above. Again when n = 2m is even, the semistable elements of X that are fixed by nontrivial connected reductive subgroups of G are those represented by polynomials such that there exist distinct p and q in P1 with exactly half the roots equal to p and the rest equal to q. They form a single Gorbit, and the stabiliser C∗ acts with weights ±4, ±6, . . . , ±n = ±2m on the normal ˜ of X this time has as its strata the to the orbit. The refined stratification {S˜β˜ : β˜ ∈ B} s set S˜(0) = X of stable points, the set S˜(T ) represented by polynomials with exactly two distinct roots each with multiplicity m = n/2, for 2 ≤ k ≤ m the set S˜(T ,2k) represented by polynomials in the orbit of one of the form am t m + am+k t m+k + am+k+1 t m+k+1 + · · · + a2m t 2m , where am and am+k are nonzero, and finally the strata S2j −n (for n/2 < j ≤ n) of the Morse stratification. Example 5.5. For a more complicated example consider the action of G = SL(3; C) and its maximal compact subgroup K = SU (3) on X = (P2 )n . A sequence (x1 , . . . , xn ) of points in P2 is semistable if and only if there is no projective line L in P2 such that |{j : xj ∈ L}| n > (5.3) 2 3 and no point p ∈ P2 such that |{j : xj = p}| >

n , 3

(5.4)

and is stable if we can replace > with ≥ in (5.3) and (5.4) (see for example [9] (16.5)). The stratification {Sβ : β ∈ B} can be described as follows (see [9] Proposition 16.9). Any (x1 , . . . , xn ) ∈ (P2 )n which is not semistable determines a unique flag 0 = M0 ⊂ M1 · · · ⊂ Ms = C3 in C3 with s = 2 or 3, such that if 1 ≤ i ≤ s, then

344

F. Kirwan

k1 ks > ··· > , m1 ms where ki = |{j : xj ∈ Mi \Mi−1 }|

and mi = dim(Mi /Mi−1 );

moreover, if mi = 2, then those xj lying in Mi \Mi−1 determine a semistable element of (P1 )ki after projection into P(Mi /Mi−1 ) ∼ = P1 . Then (x1 , . . . , xn ) lies in the stratum labelled by the projection into Lie(SU (3)) of the vector k1 ks β= ,..., ∈ Lie(U (3)) m1 ms in which each ki /mi appears mi consecutive times. Thus B is the projection into the Lie algebra Lie(SU (3)) of / n n n 0 k k 2n , , , ,n − k : 0. Note that the assertion implies all the statements of the proposition, by (2.33) and (2.34). Assume the assertion is false so that β(xψ ) = 0. But β = ψ and hence ψ − β ∈ . But then β − ψ ∈ and (β − ψ)(x−ψ ) = −2. From the representation theory of a TDS, one has that [e, [e, gβ−ψ ]] = 0. But this implies that β + ψ ∈ , contradicting the maximality of ψ.

Let ei , i = 1, . . . , d, be an orthonormal basis of gψ with respect to H|gψ . We assume that the basis is chosen so that ed = e. Under the adjoint action of uψ the element ei clearly generates a three-dimensional irreducible representation ui of uψ since [e, ei ] = 0. Of course, ud = uψ . (2.35) Remark 2.8. Note that, as a consequence of Proposition 2.7, if u=

d

(2.36)

ui ,

i=1

then u is the primary component in gC for the three-dimensional irreducible representation of uψ under the adjoint action and that any irreducible component in gC /u has dimension 1 or 2. The following lemma is well known and is readily established using the commutation relations of an S-triple. Lemma 2.9. Assume that v is a complex TDS and (x , e , f ) is an S-triple whose elements span v. Then (h, v, w) is an S-triple also spanning v, where h = i(e − f ), v = 1/2(ix + e + f ),

(2.37)

w = 1/2(−ix + e + f ). Furthermore, one recovers (x , e , f ) from (h, v, w) by x = −i(v − w), e = 1/2(−ih + v + w), f = 1/2(ih + v + w).

(2.38)

Minimal coadjoint orbits and symplectic induction

407

We apply Lemma 2.9 for the case where v = uψ and (x , e , f ) = (xψ , e, −θ e). Let h = i(e + θ e), v = 1/2(ixψ + e − θ e), w = 1/2(−ixψ + e − θ e)

(2.39)

so that (h, v, w) is an S-triple whose elements span uψ . Obviously, there exists an automorphism of uψ which carries (xψ , e, −θ e) to (h, v, w). Since any automorphism of a complex TDS is inner, it follows that xψ and h are conjugate in gC by an element in Ad(gψ )C . In particular, then, by Proposition 2.7, the multiplicity of the eigenvalue 2 of ad h in gC is d. Lemma 2.10. One has h ∈ kC so that we may write d = dk + dp ,

(2.40)

where dk is the multiplicity of the eigenvalue 2 of ad h|kC and dp is the multiplicity of the eigenvalue 2 of ad h|pC . One has dp ≥ 1. In fact, v, w ∈ pC and [h, v] = 2v. Proof. Obviously, θ h = h by (2.39) so that h ∈ kC . Similarly, v, w ∈ pC since θ v = −v and θ w = −w by (2.39), noting that xψ ∈ a ⊂ pC . One has [h, v] = 2v since (h, v, w) is an S-triple.

We can strengthen Lemma 2.10. Theorem 2.11. Let the notation be as in Lemma 2.10. Then dk = d − 1 and dp = 1. That is, the one-dimensional subspace Cv is the eigenspace of ad h|pC corresponding to the eigenvalue 2. Also 2 is the highest eigenvalue of ad h|pC . Proof. The three-dimensional uψ -modules ui (see (2.36)) are, of course, equivalent to the adjoint representation of uψ . For j = 1, . . . , d, let δj : uψ → uj be the uψ -equivalence normalized so that δj e = ej . Note that δd is the identity map. Let vj = δj v. It is then immediate from Proposition 2.7 that {vj }j = 1, . . . , d, is a basis of the ad h eigenspace in gC for the eigenvalue 2. To prove the first statement of the theorem it suffices by Lemma 2.10 to show that vj ∈ k C

for i = j, . . . , d − 1.

(2.41)

But now by the S-triple commutation relations ixψ = i[θ e, e], −θ e = −1/2[θ e, xψ ], and e = −1/2[e, xψ ]. Thus if xj , fj ∈ uj are defined by xj = [θ e, ej ] and fj = −1/2[θ e, xj ], one has (2.42) vj = 1/2(ixj + ej + fj ) by (2.39). On the other hand, [e, xj ] = [e, [θ e, ej ]] = [[e, θe], ej ] (since [e, ej ] = 0) = −[xψ , ej ] = −2ej .

(2.43)

408

B. Kostant

Let j ∈ {1, . . . , d − 1}. To establish (2.41), we will first prove that xj ∈ kC . In fact, we will prove that xj ∈ m. (2.44) Since θ|a is minus the identity, one has θ e ∈ g−ψ . But then xj clearly commutes with a. But the centralizer of a in g is m + a. To prove (2.44), it obviously suffices to prove that xj is B-orthogonal to a. But {ej , e} = {ej , ed } = 0. Thus −(ej , σu e) = −(ej , θe) = 0. But then if y ∈ a, one has (y, xj ) = (y, [θ e, ej ]) = ([ej , y], θe). But [ej , y] = −ψ(y)ej . Thus (y, xj ) = 0 establishing (2.44). To prove (2.41) it now suffices, by (2.42), to prove that θfj = ej . But θfj = −1/2[e, xj ] since θ xj = xj by (2.44). But then θfj = ej by (2.43). This proves (2.41). Since h and xψ are conjugate, the final statement of Theorem 2.11 follows from Proposition 2.7.

2.5 We retain the notation of Section 2.4, and we will the apply the results of Section 2.4 to the symplectic considerations of Section 2.2. Proposition 2.12. One has (v, w) = 1.

(2.45)

{v, v} = 1.

(2.46)

Furthermore, w = −σu v so that

Proof. Since h and xψ are conjugate, one has (h, h) = 2

(2.47)

by (2.26). But since (h, v, w) is an S-triple, one has (v, w) = 1/2([h, v], w). But ([h, v], w) = (h, [v, w]) = (h, h). Thus (2.47) implies (2.45). But now v = 1/2(ixψ + e − θ e) and w = 1/2(−ixψ + e − θ e) by (2.39). Recall σu = θ σ . But clearly σ v = 1/2(−ixψ + e − θ e) and hence θ σ v = 1/2(ixψ − e + θ e). Hence −σu v = w. But then (2.46) follows from (2.45) and (2.27).

Of course h is a hyperbolic element in kC and qh (kC ) is the parabolic subalgebra of kC defined by h. See Remark 2.2. Theorem 2.13. Under the adjoint action of kC on pC the one-dimensional subspace Cv is stable under qh (kC ). In fact, for any x ∈ qh (kC ), one has [x, v] = (h, x)v.

(2.48)

Proof. If x is contained in the nilradical of qh (kC ), then [x, v] = 0 by the last line in Theorem 2.11. On the other hand, if x ∈ (kC )h (a Levi factor of qh (kC )), then Cv is stable under ad x by the multiplicity one statement in Theorem 2.11 of the eigenvalue 2 of ad h in pC . This proves the first statement of Theorem 2.13. For x ∈ qh (kC ) let f be the linear functional on qh (kC ) defined so that [x, v] = f (x)v. But then f (x) = ([x, v], w) by (2.45). However, ([x, v], w) = (x, [v, w]) = (x, h). Thus f (x) = (h, x).


409

Let z = −ih so that z ∈ k and z = e + θ e by (2.39). Let T ⊂ K be a maximal torus such that z ∈ t. Then h ∈ h, where, as in Section 2.2, h = it. Let γ : k∗C → kC be as in (2.12), and let λ ∈ h∗ (recalling the identification h∗ = γ −1 (h)) be such that γ (λ) = h.

(2.49)

Recall that ⊂ h∗ is the T -weight lattice. Note that hC ⊂ (kC )h so that hC ⊂ qh (kC ). As an immediate consequence of Theorem 2.13, one has the following. Proposition 2.14. One has λ ∈ . Furthermore, the KC -module V generated by v with respect to the adjoint action of KC on pC is irreducible and is equivalent to Vλ with v corresponding to vλ . Henceforth we will identify V with Vλ and v with vλ . One has πλ (k)y = Ad k(y), where y ∈ V and k ∈ KC . Let ν = λ/2π i so that ν ∈ k∗ . As in Section 2.2, let X be the K-coadjoint orbit of ν so that (X, ω) is a symplectic K-homogeneous space, where ω is the KKS symplectic form. One readily notes that Lie Kν = k ∩ (kC )h

(2.50)

so that k ∩ (kC is a compact form of the Levi factor (kC of qh (kC ), where Kν is the isotropy group at ν. Furthermore, one knows (as a general fact about coadjoint orbits of compact connected Lie groups) that Kν is connected so that (2.7) and (2.8) are satisfied, where χ is the character on Kν defined by the action of Kν on Cvλ . Thus ωX as in Section 2.2, we can construct the induced symplectic manifold (X, ). As in Section 2.2 let E ⊂ Vλ be the variety of extremal weight vectors so that E = πλ (KC )C∗ vλ . Let Hλ be the K-invariant Hilbert space structure in Vλ given the restriction H|Vλ . As in Section 2.2, E 1 is the space of vectors in E having length 1 with respect to Hλ . Note that vλ ∈ E 1 (2.51) )h

)h

by (2.46). We recall that Proposition 2.3 sets up a K × U (1) isomorphism L1 → E 1

(2.52)

→E X

(2.53)

and a K × U (1) × R+ isomorphism

Let Kv be the isotropy group at v = vλ for the action of K on E 1 and let Ke be the isotropy group at e ∈ g for the adjoint action of K on g. Theorem 2.15. The following three subgroups of K are equal: (1) Kv ; (2) Ke ; (3) the centralizer of the TDS uλ in K.

410

B. Kostant

Proof. Let K be the subgroup of K defined by (3). Since v, e ∈ uψ , one obviously has K ⊂ Kv and K ⊂ Ke . But clearly Ad k commutes with θ for any k ∈ K. Thus θ (e) is fixed by Ad k for any k ∈ Ke . But then all three elements of the S-triple in Proposition 2.6 are fixed by Ad k. Hence Ke = K by the definition of uψ (see Section 2.3). But σu also commutes with the adjoint action of K since k ⊂ gu . But w = −σu v by Proposition 2.12. Thus w is fixed by Ad k for any k ∈ Kv . Hence any such k fixes the three elements of the S-triple (h, v, w). But these elements also span uψ . Thus K = Kv .

Let O be the Ad G orbit of e in g and let O 1 = {f ∈ O | {f, f } = 1}. Note that e ∈ O 1 by the choice of e in Section 2.3. Since K operates unitarily with respect to H, the adjoint action of k stabilizes E 1 and O 1 . As a corollary of Theorem 2.15, one has the following. Theorem 2.16. The compact group K operates transitively on E 1 and on O 1 . Furthermore, these spaces are isomorphic as K-homogeneous spaces. In fact, b is such an isomorphism, where for any k ∈ K, b(Ad k(vλ )) = Ad k(e).

(2.54)

Proof. Recall that z = e + θ e = −ih ∈ k. But if s ∈ R, one has πλ (exp sz)vλ = e−2si vλ

(2.55)

by (2.47) and (2.48). In particular, k → φ(k, 1) in (2.19) surjects k onto E 1 by Proposition 2.3. Consequently, K operates transitively on E 1 . On the other hand, if A and N are the subgroups of G which correspond, respectively, to a and n then one has the group Iwasawa decomposition G = KAN . But e is fixed under the adjoint action of N since e ∈ Cent n (see Proposition 2.5). On the other hand, Ad A(e) = R+ e. Thus O = Ad KR+ e. (2.56) However, clearly R+ e∩O 1 = {e}. Hence K operates transitively on O 1 . The theorem then follows from the equality of (1) and (2) in Theorem 2.15.

The variety E is KC homogeneous by Remark 2.4. The KC orbit E in pC corresponds to the G-orbit O in g by the Kostant–Sekiguchi correspondence (a correspondence of KC nilpotent orbits in pC and G nilpotent orbits in g; see [S]). Michèle Vergne has proved the corresponding orbits are K-diffeomorphisms (see [V]). The proof is highly nontrivial. However, by Theorem 2.16, in the special case of E and O the diffeomorphism is transparent. Obviously, by (2.21) and (2.56), one has K × R+ diffeomorphisms E 1 × R+ → E, (f, t) → tf, (2.57) 1 + (u, t) → tu. O × R → O, We may therefore extend the domain of definition of b so that, using the notation of (2.57), one has a K × R+ -diffeomorphism b : E → O,

where b(tf ) = tb(f ).

(2.58)


411

ω ) ∼ 3 The symplectic isomorphism (X, X = (Z, ωZ ) 3.1 We continue with the notation of Section 2. Recalling (2.12), one notes that since Bk = B|kC and since kC and pC are B-orthogonal, the isomorphism g∗C to gC defined by B is an extension of (2.12). The extension will also be denoted γ . Let ε ∈ g∗ be defined so that γ (ε) = e/π. (3.1) Let Z ⊂ g∗ be the G-coadjoint orbit of ε and let ωZ be the KKS-symplectic form on Z. To avoid confusion with the vector field ξ x on X (see Section 2.1) defined by any x ∈ k, with respect to the coadjoint action of K on X, we will denote by +y the vector field on Z defined by any y ∈ g with respect to the coadjoint action of G on Z. The analogue of (2.2) is the formula ωZ (+x , +y )(ρ) = ρ, [y, x]

(3.2)

for any ρ ∈ Z. In particular, if ρ = ε, one has ωZ (+x , +y )(ε) = (1/π)(e, [y, x]).

(3.3)

Recall that ω is the KKS form on the K-coadjoint orbit X of ν = λ/2π i. Lemma 3.1. Let x, y ∈ k. Then ωZ (+x , +y )(ε) = ω(ξ x , ξ y )(ν).

(3.4)

Proof. [y, x] is fixed by θ since [y, x] ∈ k. Thus (1/π )(e, [y, x]) = ((e + θ e)/2π, [y, x]). But e + θ e = (1/ i)h by (2.39) and γ (λ) = h. But then γ (ν) = (e + θ e)/2π.

(3.5)

Thus (1/π )(e, [y, x]) = ν, [y, x]. But then (3.4) follows from (2.2) and (3.3).

Now recalling (2.9), the circle bundle L1 is given by L1 = K ×Kν U (1), where the action of Kν on U (1) is given by the character (recall that Kν is connected) χ (exp x) = eλ(x) = e(h,x)

(3.6)

= L1 × R+ so that for any x ∈ kν (see (2.48)). Now by (1.17) one has X = K ×Kν U (1) × R+ . X

(3.7)

be the point whose components are the identity in K, 1 in U (1), and 1 in Let o ∈ X + R with respect to (3.7). Extend the domain of the bundle projection τ (see (1.6)) to so that τ (q, t) = τ (q) for (q, t) ∈ L1 × R+ . One notes that X τ (o) = ν.

(3.8)

412

B. Kostant

Proposition 3.2. There exists a K × R+ diffeomorphism → Z, β:X

(3.9)

β(tk · o) = t (Coad k(ε)).

(3.10)

where . The result then follows from Proposition 2.3, Proof. Put β = (1/π )γ −1 ◦ b ◦ φ Theorem 2.16, (2.58), and the invariance of B.

3.2 ωX Our main objective will be to prove that β : (X, ) → (Z, ωZ ) is an isomorphism of symplectic manifolds. → T (Z) be the diffeomorphism of tangent bundles defined by the Let β∗ : T (X) so that differential of β. Let βo be the restriction of β∗ to the tangent space To (X) → Tε (Z) βo : To (X)

(3.11)

defined by the is a linear isomorphism. For any x ∈ k, let ηx be the vector field on X Since β is a K-map, one has action of K on X. β∗ (ηx ) = +x .

(3.12)

One can be very explicit about ηx . Proposition 3.3. Let x ∈ k. Then using the notation of (1.13) and (2.4), one has Gx ζ. ηx = ξx + ϕ

(3.13)

ηx is characterized by the property Proof. As a vector field on L1 (and hence on X), that (1) it commutes with the U (1)-action, (2) it annihilates α by Lie differentiation, and (3) τ∗ (ηx ) = ξ x . (3.14) The result then follows from (1.13), (2.5), and Theorem 1.2.

Let k⊥ ν be the B-orthocomplement of kν in k so that the map k⊥ ν → Tν (X)

(3.15)

given by x → (ξ x )ν is a linear isomorphism. Let Ro be the space of horizontal tangent vectors (i.e., orthogonal to α) to L1 at o so that Ro has codimension 1 in To (L1 ) and codimension 2 in To (X). Lemma 3.4. One has (ηx )o ∈ Ro for any x ∈ k⊥ ν and the map k⊥ ν → Ro , is a linear isomorphism.

x → (ηx )o

(3.16)


413

Proof. Let x ∈ kν⊥ . Then ϕ x (ν) = 0 by (2.4) since γ (ν) ∈ kν . Thus (ηx )o = ξx

(3.17)

by (3.13). This proves that (ηx )o ∈ Ro . But since τ∗ : Ro → Tν (X) is clearly an isomorphism the remaining statements of the proposition follow from (3.14) and the isomorphism (3.15).

Let Rε = βo (Ro ) so that (3.11) restricts to the linear isomorphism βo : Ro → Rε . induced by the retriction of ωX Let ωo be the symplectic bilinear form on To (X) to To (X), and let ωε be the symplectic bilinear form on Tε (Z) induced by the retriction of ωZ to Tε (Z). We wish to prove that βo : (To (X), ωo ) → (Tε (Z), ωε )

(3.18)

is an isomorphism of symplectic vector spaces. We first establish the following. Lemma 3.5. The restrictions ωo |Ro and ωε |Rε are nonsingular and βo : (Ro , ωo |Ro ) → (Rε , ωε |Rε )

(3.19)

is an isomorphism of symplectic vector subspaces. ⊥ Proof. Recalling the definition of ωX (see (1.19)) it is clear that if x, y ∈ kν , then x y x y x y x y ωX ω(ξ , ξ )(o) by (3.17). But ωX (η , η )(o) = (η , η )(o) = ω(ξ , ξ )(ν). Thus ωo |Ro is nonsingular by the linear isomorphism (3.15). But then ωε |Rε is nonsingular and (3.19) is an isomorphism of symplectic vector subspaces by (3.4) and (3.12).

with respect Now let Ro⊥ be the two-dimensional orthocomplement of Ro in To (X) to ωo . It is clear from (1.19) and Section 1.2 that Ro⊥ is spanned by ζo and (d/dr)o . It will be convenient for us to modify this basis of Ro⊥ . Recall that z ∈ k is given by z = e + θ e. Lemma 3.6. One has (ηz )o = −ζo /π so that

(ηz )

o

and (−2rd/dr)o are a basis of

Ro⊥ .

(3.20) Furthermore,

ωo ((−2rd/dr)o , (ηz )o ) = −2/π.

(3.21)

Proof. By (2.49) one has γ (ν) = z/2π (3.22) z z z ζ )o by (3.13). But ϕ (o) = ϕ z (ν) so that z ∈ kν . Thus ν = 0. Hence (η )o = (ϕ z z and ϕ (ν) = (γ (ν), z) by (2.4). Hence ϕ (o) = 1/2π(z, z) by (3.22). But since z = −ih one has (z, z) = −2 by (2.47). This proves (3.20). But now by (1.19), since r(o) = 1, (ξ z )

ωo ((−2rd/dr)o , (ηz )o ) = (dr ∧ α)(−2rd/dr, ηz )(o) = −2/π by (3.20) and (1.10). This proves (3.21).

414

B. Kostant

Let κ be the Euler vector field on Z. Thus if f ∈ C ∞ (Z) and µ ∈ Z, then (κf )(µ) = d/dtf (µ + tµ)|t=0 . Clearly, β∗ (rd/dr) = κ.

(3.23)

βo ((−2rd/dr)o ) = (+xψ )ε

(3.24)

Lemma 3.7. One has (see Proposition 2.6). Proof. One has [xψ , e] = 2e by Proposition 2.6. But then coad xψ (ε) = 2ε

(3.25)

since π γ is an equivalence of g-modules (see (3.1)). But (+xψ )ε = −2κε . (See the beginning of Section 2.1 to explain the minus sign.) But then (3.24) follows from (3.23).

Lemma 3.8. One has ωε ((+xψ )ε , (+z )ε ) = −2/π.

(3.26)

Proof. ωε ((+xψ )ε , (+z )ε ) = ωZ (+xψ , +z )(ε) = ε, [z, xψ ] = (1/π)(e, [z, xψ ]) = (1/π)([e, e + θ e], xψ ) = −(1/π)(xψ , xψ ) = −2/π

by Proposition 2.6

by (2.26).

We can now prove the following. Theorem 3.9. The map βo : (To (X), ωo ) → (Tε (Z), ωε )

(3.27)

is an isomorphism of symplectic vector spaces. Proof. Let Rε⊥ be the two-dimensional orthocomplement of Rε in Tε (Z) with respect to ωε . We assert (Assertion A) that (+z )ε and (+xψ )ε is a basis of Rε⊥ . We first show that (+z )ε ∈ Rε⊥ . To do this it suffices to show that ωZ (+z , +x )(ε) = 0

(3.28)

for all x ∈ k since Rε is spanned by (+x )ε for x ∈ k⊥ ν , by Lemmas 3.4 and 3.5. But if x ∈ k, then ωZ (+z , +x )(ε) = 1/π(e, [x, z])


415

= (1/2π)((e + θ e), [x, z]) since [x, z] ∈ k = (1/2π )([z, z], x) = 0. Thus (+z )ε ∈ Rε⊥ . Let y ∈ k⊥ ν . Then ωZ (+xψ , +y )(ε) = (1/π)(e, [y, xψ ]) = (1/π)([xψ , e], y) = (2/π)(e, y) by Proposition 2.6 = (1/π)(e + θ e, y) since y ∈ k = 0 since z ∈ kν and y ∈ k⊥ ν. But then (+xψ )ε ∈ Rε⊥ by Lemmas 3.4 and 3.5. This proves Assertion A since the left side of (3.26) is nonzero. But now we assert (Assertion B) that βo (Ro⊥ ) ⊂ Rε⊥ and βo : (Ro⊥ , ωo |Ro⊥ ) → (Rε⊥ , ωε |Rε⊥ )

(3.29)

is an isomorphism of symplectic subspaces. Indeed, βo ((ηz )o ) = (+z )ε by (3.12) and βo ((−2rd/dr)o ) = (+zψ )ε by (3.24). But then Assertion B follows from Assertion A together with Lemma 3.6 and the fact that −2/π occurs on the right side of (3.21) and on the right side of (3.26). But then the theorem follows from the symplectic isomorphism (3.29) together with the symplectic isomorphism (3.19).

The following is our main result. Theorem 3.10. Let G be a connected noncompact Lie group with finite center such that Lie g is simple. Let K be a maximal compact subgroup and let X be the coadjoint ωX orbit of K defined as in Section 2.5. Let (X, ) be the symplectic manifold obtained = dim X + 2. See Section 1.3. Let from X by symplectic induction so that dim X (Z, ωZ ) be the coadjoint orbit of G, together with its KKS symplectic form, defined as in Section 3.1, and let ωX β : (X, (3.30) ) → (Z, ωZ ) be the K-diffeomorphism (a special case of M. Vergne’s theorem) defined as in Section 3.1 using the Kostant–Sekiguchi correspondence. Then (3.30) is an isomorphism of symplectic manifolds. Proof. Note that L1 (see (2.9)) is K-homogeneous since (2.7) is surjective (ν = 0 is K × R+ homogeneous by (1.17). For any (k, s) ∈ since G is noncompact). Thus X + defined by the action of (k, s) on X. K × R , let k,s be the diffeomorphism of X Thus if q ∈ X, then k,s (q) = s(k · q). Let mk,s be the diffeomorphism of Z defined so that if µ ∈ Z, then mk,s (µ) = s(Coad k(µ)). It follows from (2.56) that O is K × R+ homogeneous. Consequently, Z is K × R+ homogeneous since (see (3.1)) π γ : Z → O obviously commutes with the action of K × R+ . From the definition of β (see (3.10)), it is immediate that one has the commutative diagram equality of maps

416

B. Kostant

β ◦ k,s = mk,s ◦ β.

(3.31)

and put p = k,s q. We assert that the pullback Let q ∈ X (k,s )∗ ((ωX )p ) = s(ωX )q .

(3.32)

But recalling (1.19), it is obvious that α and ω are invariant under k,s . On the other hand, clearly (k,s )∗ r = sr and hence (k,s )∗ dr = sdr. This proves (3.32). Now let µ ∈ Z and let ρ = mk,s (µ). We assert that (mk,s )∗ ((ωZ )ρ ) = s(ωZ )µ .

(3.33)

Since ωZ is obviously K-invariant it suffices to prove (3.33) under the assumption that k is the identity of K. Making that assumption, one has ρ = sµ. But also +y for any y ∈ g is invariant under mk,s . Thus for any y ∈ g, one has (mk,s )∗ ((+y )µ ) = (+y )sµ .

(3.34)

But then for any x, y ∈ g, one has (mk,s )∗ ((ωZ )sµ )((+x )µ , (+y )µ ) = (ωZ )sµ ((+x )sµ , (+y )sµ ) = sµ, [y, x] = s(ωZ )µ ((+x )µ , (+y )µ ). be arbitrary and let µ = βp. To prove Theorem 3.10, But this proves (3.33). Let p ∈ X it suffices to show that β ∗ ((ωZ )µ ) = (ωX (3.35) )p . By transitivity, there exists (k, s) ∈ K × R+ such that k,s p = o. But then mk,s µ = ε by the commutativity equation (3.31) and, in fact, β ∗ ((ωZ )µ ) = (k,s )∗ ((βo )∗ (((mk,s )−1 )∗ (ωZ )µ )). However, (mk,s )−1 )∗ (ωZ )µ = s −1 (ωZ )ε by (3.33). But (βo )∗ (s −1 (ωZ )ε ) = s −1 (ωX )o by Theorem 3.9. Finally, (k,s )∗ (s −1 (ωX ) ) = (ω ) by (3.32). This proves o p X (3.35).

3.3 We wish to characterize the varieties Z and X in more general terms. Recall (E. Cartan’s theory) that the noncompact symmetric space G/K is one of two types: (1) nonHermitian symmetric or (2) Hermitian symmetric. In the non-Hermitian case, pC is KC -irreducible and kC is semisimple. In the Hermitian case, Cent kC is one dimensional and if I is a set indexing the KC -irreducible submodules V i , i ∈ I , of pC , then I is a two-element set and pC = V i. (3.36) i∈I

Also, if i ∈ I , there exists a linear isomorphism δi : Cent kC → C such that V i = {u ∈ pC | ad x(u) = δi (x)u ∀x ∈ Cent kC }. In addition, one has

(3.37)


δi = −δi ,

417

(3.38)

{i, i }

where = I. In case (1), we will say that g is of non-Hermitian type, and in case (2), we will say that g is of Hermitian type, Recall that gψ = Cent n, and we have put d = dim gψ . See Sections 2.3 and 2.4. Proposition 3.11. If d > 1, then M is transitive on the unit sphere S (relative to H) in gψ . Furthermore, g is of Hermitian type if and only if (a) d = 1 and (b) M operates trivially on gψ . Proof. The transitivity statement actually is stated in [K-2, Theorem 2.1.7 and the remark that follows it]. However, one need not use that reference. We have already established what is needed to prove transitivity on S in the present paper. Indeed, by (2.43) and (2.44), one has that [m, e] spans the H orthocomplement of Re in gψ . This implies Ad M(e) is open in S. On the other hand, it is also closed since M is compact. Thus Ad M(e) = S if d > 1 since S is connected if d > 1. In any case, one has Ad G(e) = Ad K(R+ e) (3.39) by the Iwasawa decomposition G = KAN . But Ad G(e) and hence also Ad K(e) spans g by the simplicity of g. But if g is of Hermitian type, then certainly Cent k = 0 and if 0 = x ∈ Cent k the function f (k) = (Ad k(e), x) on K is constant, real, and nonzero. But then −e ∈ / Ad Me. Hence d = 1 and M operates trivially on gψ by the transitivity statement. Conversely, if d = 1 and M operates trivially on gψ , then the line Ce is stable under the complex parabolic subalgebra (m + a + n)C . But then e generates a complex irreducible ad gC -module, necessarily containing g, and hence equal to gC . Thus gC is simple and e is the extremal weight vector corresponding to (m + a + n)C . But then gC is a spherical ad gC -module by the Cartan–Helgason theorem. Any nonzero spherical vector must clearly lie in kC (e.g., by (3.37), (3.38), and the simplicity of gC ). But then Cent kC = 0. Thus g is of Hermitian type.

Remark 3.12. Note that as a consequence of Proposition 3.11, one has the statement −e ∈ / Ad M(e) ⇐⇒ g is of Hermitian type.

(3.40)

But one also has the statement −e ∈ / Ad G(e) ⇐⇒ g is of Hermitian type.

(3.41)

Indeed, if g is of non-Hermitian type, then −e ∈ Ad M(e) by (3.40) and hence, of course, −e ∈ Ad G(e). If g is of Hermitian type, let 0 = x ∈ Cent k. If −e ∈ Ad G(e), then the function f in the proof of Proposition 3.11 must change signs by (3.39) and hence cannot be constant. This proves (3.41). Let Proj(g∗ ) be the real projective space defined by g∗ and let P : g∗ − {0} → Proj(g∗ ) be the projectivization map. Let C = γ −1 (Cent n) so that ε ∈ C ⊂ g∗ (see Proposition 2.5 and (3.1)).

418

B. Kostant

= in Proj(g∗ ) so that if Y = is any Theorem 3.13. There exists a unique closed G-orbit Z ∗ = = G-orbit in Proj(g ), then Z is contained in the closure of Y . In particular, = ≥ dim Z = dim Y

(3.42)

= = Z. = and equality occurs in (3.41) if and only if Y ∗ = if Furthermore, if Z ⊂ g is any nonzero G-coadjoint orbit, then Z ⊂ P −1 (Z) and only if Z is of the form Coad G(e ) for e ∈ C − {0}. In fact, using the notation of Theorem 3.10, one has = Z = P −1 (Z) (3.43) in case g is of non-Hermitian type. In particular, Z = −Z in the non-Hermitian case. If g is of Hermitian type, let J be an index set parameterizing all G-coadjoint orbits, = Then J is a two-element set and one has Z j , j ∈ J , in P −1 (Z). {Z, −Z} = {Z j },

j ∈ J,

(3.44)

so that Z = −Z in the Hermitian case. In either case, one has dim Y ≥ dim Z

(3.45)

for any nonzero coadjoint G-orbit Y . Proof. Let 0 = x ∈ g. Then the span g1 of Ad g(x) over all g ∈ G is a nonzero ideal in g and hence g1 = g. Thus there exists g ∈ G such that the component x of Ad g(x) in gψ with respect to the decomposition g=m+a+

gϕ ϕ∈

is not zero. But then by Proposition 2.7, one has lim P (Ad(exp txψ )(x)) = P (x ),

t→+∞

(3.46)

where we also let P denote the projection map of g onto Proj(g). On the other hand, if x ∈ gψ − {0}, then P (Ad G(x )) = P (Ad G(x )) by Proposition 3.11. But P (Ad G(x )) is compact since P (x ) is fixed by the action of AN and hence P (Ad G(x )) = K · P (x ). But P −1 (P (Ad G(x )) is a single Ad G-orbit by Proposition 3.11 and (3.40) in case g is of non-Hermitian type. On the other hand, it decomposes into a union of two distinct Ad G orbits, one the negative of the other, by Proposition 3.11 and (3.41), in case g is of Hermitian type. Since γ : g∗ → g is a

G-equivalence the statements above clearly carry over to g∗ . Remark 3.14. Because g is simple and Z is a G-coadjoint orbit there exists a Lie algebra injective homomorphism g → C ∞ (Z) (of course, with respect to the Poisson algebra structure on C ∞ (Z)). But then the symplectic isomorphism (3.30) implies that there exists a Lie algebra injective homomorphism


419

g → C ∞ (X). is the smallest By the coadjoint orbit covering theorem and (3.45) note that dim X possible dimension of a symplectic manifold W which admits an embedding of g as a Lie algebra of functions on W under Poisson bracket. This points to an interesting ωX difference between (X, ω) and the induced symplectic manifold (X, ) in that one cannot have a nontrivial Lie algebra homomorphism g → C ∞ (X) since dim X = dim Z − 2

(3.47)

by (1.18). If V is a complex finite-dimensional irreducible K (and hence KC module), let X(V ) ⊂ k∗ be the integral K-coadjoint orbit associated to V by the Borel– Weil theorem. Thus if v ∈ V is an extremal weight vector there exists a Cartan subalgebra hC of kC , which is the complexification of a Cartan subalgebra of k, such that v is an hC -weight vector for an extremal hC -weight λ. We may regard λ ∈ k∗C , where λ|[hC , kC ] = 0. Then ν = λ/2π i is real on k and X(V ) is the coadjoint orbit of ν. It is straightforward to show that X(V ) is independent of the choice of hC . The embedding k → g induces, by transpose, a surjection µg,k : g∗ → k∗ .

(3.48)

Remark 3.15. Note that if Y is a G-coadjoint orbit, then the restriction µg,k |Y is the moment map for the action of K on (Y, ωY ), where ωY is the KKS-symplectic form on Y . Indeed, this follows immediately from (2.4), where G replaces K and Y replaces X. Theorem 3.16. We use the notation of Theorem 3.10. One has µg,k (Z) = R+ X.

(3.49)

Moreover, if g is of non-Hermitian type, then X = X(pC ). Also, X = −X in the non-Hermitian case. If g is of Hermitian type, let X i = X(V i ) for i ∈ I (see (3.37)). Then X = −X and {X, −X} = {X i }, i ∈ I. (3.50) Furthermore (recalling (3.44)), there exists a unique bijection α : I → J such that for i ∈ I , (3.51) µg,k (Z α(i) ) = R+ X i . If X = Xi , then Z = Z α(i) . Finally, adding to the symplectic isomorphism (3.30), for any i ∈ I , there exists a symplectic K-diffeomorphism Gi , ωG ) → (Z α(i) , ω α(i) ), βi : (X Z Xi where ωZ α(i) is the KKS form on the G-coadjoint orbit Z α(i) .

(3.52)

420

B. Kostant

Proof. Let p : g → k be the projection corresponding to the Cartan decomposition g = k + p. Obviously, p ◦ γ = γ ◦ µg,k (3.53) on g∗ . Recall (see Section 2.5) that O is the G-adjoint orbit of e. But O = Ad KR+ e by (2.56). Thus f ∈ O if and only if there exists t ∈ R+ and k ∈ K such that f = t Ad k(e/π). But clearly p(e/π) = (e + θe)/(2π ). That is p(e/π ) = h/(2π i) by (2.39). Thus p(f ) = t Ad k(h/(2π i)). Applying γ −1 to both sides, one has µg,k (γ −1 (f )) = t Coad k(γ −1 (h)/(2π i)) by (3.53). But O = γ (Z) (see Section 3.1) so that if ρ = γ −1 (f ), then ρ ∈ Z and the most general element in Z is of this form. Furthermore, γ −1 (h) = λ (see (2.49)) and ν = λ/(2π i) (see Section 2.5). Thus µg,k (ρ) = t Coad k(ν)). Since k ∈ K and t ∈ R+ are arbitrary and X is the K-coadjoint orbit of ν, this proves (3.49). Now since B|pC is nonsingular, it follows that pC as a K-module is selfcontragedient. In particular, µ is a weight of pC ⇐⇒ −µ is a weight of pC .

(3.54)

Recall the choice of X in Section 2.5. By definition X = X(Vλ ),

(3.55)

where Vλ is the K-irreducible submodule of pC defined in Section 2.5 with extremal weight vector v (see (2.48)). Assume g is of non-Hermitian type. Then pC is Kirreducible so that Vλ = pC . This proves X = X(pC ). But then X = −X by (3.54). Now assume that g is of Hermitian type. Then Vλ = V i for some i ∈ I . But µ| Cent k = δi | Cent k for any weight µ of Vλ by (3.37). Thus X = −X and one easily has (3.50) by (3.54). But (3.49) implies µg,k (−X) = R+ (−Z). But then (3.51) follows from (3.44) and (3.49). The choice of e ∈ gψ was arbitrary (see Section 2.3) subject only to the condition that {e, e} = 1. We can therefore replace e by −e. In that case h would be replaced by −h and λ by −λ. Consequently, X is replaced by −X and Z by −Z. Thus the argument which leads to the symplectic K-isomorphism (3.30) yields a symplectic C ω−X K-diffeomorphism (−X,

C ) → (−Z, ω−Z ). This implies (3.52). 3.4 Even though g is simple the complexification gC may not be simple. Indeed, this is the case if g itself were complex but its complex structure is ignored. We will say that g is Omin -split if gC is a simple complex Lie algebra and e ∈ Omin , where Omin is the minimal nilpotent orbit in gC . Note that by the transitivity statement in Proposition 3.11 and Theorem 3.13, the definition of Omin -split depends only on g and is, in particular, independent of the choice of e. If g is Omin -split, then dim Z = 2h∨ − 2,

(3.56)


421

where h∨ is the dual Coxeter number of gC . This is clear since one knows dimC Omin = 2h∨ − 2. But by the irreducibility of the adjoint representation of gC one has Omin = Ad gC (e). However, O = Ad g(e) (see Section 2.5). But then (3.56) follows by computing the dimension of the respective tangent spaces at e. See Section 3.1 for the definition of Z. Theorem 3.17. The simple Lie algebra g is Omin -split if and only if dim Cent n = 1.

(3.57)

Proof. If dim Cent n = 1 then Ce is stabilized, under the adjoint represention, by the complex parabolic subalgebra (m + a + n)C . But then e generates an irreducible gC -module under the adjoint representation of gC . But this module contains g by the simplicity of g. Hence the module equals gC so that gC is simple. Furthermore, e ∈ Omin since e is an extremal weight vector of this module. Thus g is Omin -split. Conversely assume that g is Omin -split. Then uψ (see Section 2.3) is conjugate to the TDS of a highest root vector in gC by [K-3, Corollary 3.6]. Since the root in question is long, the multiplicity of the eigenvalue 2 of ad xψ is 1. Thus d = 1 by Proposition 2.7. That is, dim Cent n = 1. See Section 2.4.

Examples 3.18. By Theorem 3.17, g is Omin -split if (a) g is split (so that all restricted root spaces are one dimensional); (b) gC is simple and g is a quasi-split form of gC (since nC is a maximal nilpotent Lie algebra of gC ); (c) g is of Hermitian type (by Proposition 3.11). Note that if g is Omin -split, then dim X = 2h∨ − 4

(3.58)

by (3.47) and (3.56). In general, X ∼ = K/Kν can be given the structure of a partial complex flag manifold (see (2.16)). If g is Omin -split, much more can be said. Proposition 3.19. If g is Omin -split (e.g., if g is split), then X is not only a Ksymmetric space but, in fact, X is a Hermitian symmetric space. Proof. Recall the notation of Section 2.4. If g is Omin -split then by Theorem 3.17 the number dk in Theorem 2.11 is 0. Thus since xψ and h are conjugate, the eigenvalues of ad h|kC are in the set {1, 0, −1}. Since (kν )C is the ad h|kC -eigenspace for the eigenvalue 0 the result is immediate.

Remark 3.20. Assume that g is Omin -split and g is of non-Hermitian type so that kC is semisimple. Let K be a noncompact real form of KC having Kν as a maximal compact subgroup so that K /Kν = X is the noncompact symmetric dual to the compact symmetric space X. But now X = −X by Theorem 3.16 so that h and −h are K-conjugate. One readily shows that this implies that h lies in a TDS of kC so that not only is X a complex bounded domain but, in fact, X is a tube domain. See [K-W]. In particular, by the Kantor–Koecher–Tits theory, X corresponds to a formally real

422

B. Kostant

Jordan algebra J (X). See [K-S, Section 5] for a classification of the simple formally real Jordan algebras and the corresponding tube domains. One then has dim X = 2 dim J (X).

(3.59)

If g is a split form of any one of five exceptional simple Lie algebras, g is nonHermitian so that Remark 3.20 applies to g. But a minimal (dimensional) symplectic realization of g as functions on a symplectic manifold is achieved when the man of a coadjoint orbit of a compact Lie group K. ifold is the induced symplectic X See Remark 3.14. The group K turns out to be classical in all five cases so that the exceptional Lie algebras g emerge symplectically from the symplectic induction of a classical coadjoint orbit. The table below contains the relevant information. The cases of E6 , E7 , and E8 are taken from [B-K]. To avoid complicated notation, the compact groups listed below are correct only up to finite coverings. The symbol H (n)/F denotes the Jordan algebra of n × n Hermitian matrices over the field F . The compact form of Sp(2n, C) will be denoted simply by Sp(2n). gC type K X dim X J (X) G2 SU (2) × SU (2) P1 (C) × P1 (C) 4 R⊕R F4 SU (2) × Sp(6) P1 (C) × (Sp(6)/U (3)) 14 R ⊕ (H (3)/R) E6 Sp(8) Sp(8)/U (4) 20 H (4)/R SU (8) SU (8)/(SU (4) × SU (4) × U (1)) 32 H (4)/C E7 E8 Spin(16) Spin(16)/U (8) 56 H (4)/H

References [B-K] R. Brylinski and B. Kostant, Lagrangian models of minimal representations of E6 , E7 , and E8 , in S. Gindikin, J. Lepowsky, and R. L. Wilson, eds., Functional Analysis on the Eve of the 21st Century: In Honor of the Eightieth Birthday of I. M. Gelfand , Progress in Mathematics, Vol. 131, Birkhäuser, Boston, 1995, 13–53. [K-1] B. Kostant, Quantization and unitary representations, in C. T. Taam, ed., Lectures in Modern Analysis III, Lecture Notes in Mathematics, Vol. 170, Springer-Verlag, New York, 1970, 87–207. [K-2] B. Kostant, On the existence and irreducibility of certain series of representations, in I. M. Gelfand, ed., Lie groups and Their Representations, Wiley, New York, 1971, 231–329. [K-3] B. Kostant, The principal three-dimensional subgroup and the Betti numbers of a complex simple Lie group, Amer. J. Math., 81-4 (1959), 973–1032. [K-S] B. Kostant and S. Sahi, The Capelli identity, tube domains, and the generalized Laplace transform, Adv. Math., 87 (1991), 71–92. [K-W] A. Koranyi and J. Wolf, Realization of Hermitian symmetric spaces as generalized half-planes, Ann. Math., 81 (1965), 265–288. [S] J. Sekiguchi, Remarks on real nilpotent orbits of a symmetric pair, J. Math. Soc. Japan, 39 (1987), 127–138. [V] M. Vergne, Instantons et correspondance de Kostant–Sekiguchi, C. R. Acad. Sci. Paris Sér. I Math., 320 (1995), 901–906.

Quantization of pre-quasi-symplectic groupoids and their Hamiltonian spaces∗ Camille Laurent-Gengoux and Ping Xu Department of Mathematics Pennsylvania State University University Park, PA 16802 USA [email protected], [email protected] Dedicated to Alan Weinstein on the occasion of his 60th birthday. Abstract. We study the prequantization of pre-quasi-symplectic groupoids and their Hamiltonian spaces using S 1 -gerbes. We give a geometric description of the integrality condition. As an application, we study the prequantization of the quasi-Hamiltonian G-spaces of Alekseev– Malkin–Meinrenken.

1 Introduction Quasi-symplectic groupoids are natural generalizations of symplectic groupoids [7, 22]. The main motivation of [22] in studying quasi-symplectic groupoids was to introduce a single, unified momentum map theory in which ordinary Hamiltonian G-spaces, Lu’s momentum maps of Poisson group actions, and the group-valued momentum maps of Alekseev–Malkin–Meinrenken can be understood under a uniform framework. An important feature of this unified theory is that it allows one to understand the diverse theories in such a way that techniques in one can be applied to the others. It turns out that much of the theory of Hamiltonian spaces of a symplectic groupoid can be generalized to quasi-symplectic groupoids. In particular, one can perform reduction and prove that J −1 (O)/ is a symplectic manifold, where O ⊂ M is an orbit of the groupoid ⇒ M. More generally, one can introduce the classical intertwiner space X2 × X1 between two Hamiltonian -spaces X1 and X2 , generalizing the notion studied by Guillemin–Sternberg [10] for ordinary Hamiltonian G-spaces. One shows that this is a symplectic manifold (whenever it is a smooth manifold). In particular, when is the AMM quasi-symplectic groupoid [6, 22], this reduced space describes the symplectic structure on the moduli space of flat connections on a surface [3]. ∗ This research was partially supported by NSF grant DMS03-06665.

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C. Laurent-Gengoux and P. Xu

As in the case of symplectic groupoids [20], one can introduce Morita equivalence for quasi-symplectic groupoids. In particular, it has been proved [22] that (i) Morita-equivalent quasi-symplectic groupoids give rise to equivalent momentum map theories in the sense that there is a bijection between their Hamiltonian spaces; (ii) the classical intertwiner space X2 × X1 is independent of the Morita equivalence class of . This Morita invariance principle accounts for various well-known results concerning the equivalence of momentum maps, including the Alekseev–Ginzburg– Weinstein linearization theorem [1, 9] and the Alekseev–Malkin–Meinrenken equivalence theorem for group-valued momentum maps [3] (see [22] for details). One important feature of Hamiltonian G-spaces is the Guillemin–Sternberg theorem which states that “[Q, R] = 0’’: quantization commutes with reduction [10, 13]. One expects that “[Q, R] = 0’’ should be a general guiding principle for all momentum map theories. To carry out such a quantization program, the first important step is the construction of prequantum line bundles. In this paper, we study the prequantization of Hamiltonian spaces for quasi-symplectic groupoids. Our method uses the theory of S 1 -bundles and S 1 -gerbes over a groupoid along with their characteristic classes, as developed in [4, 5]. Roughly, our construction can be described as follows. Aprequantization of a quasi-symplectic groupoid ( ⇒ M, ω+ ) is an S 1 -central extension R → of the groupoid ⇒ M (or an S 1 -gerbe over the groupoid) equipped with a pseudo-connection having ω + as pseudo-curvature. Such a prequantization exists if and only if ω + is a de Rham integral 3-cocycle and is exact (assuming that is a proper groupoid). A prequantization of a Hamiltonian space is then an S 1 -bundle L over R ⇒ M together with a compatible pseudo-connection, where the R-action on L is S 1 -equivariant. A prequantization of the symplectic intertwiner space X2 × X1 can be constructed using these data. Indeed one can show that R\(L1 ×M L2 ) is a prequantization of the symplectic intertwiner space X2 × X1 , and the natural 1-form on L1 ×M L2 induced by the connection forms on L1 and L2 descends to a prequantization connection on the quotient space R\(L1 ×M L2 ). When is not exact, one must pass to a Morita-equivalent quasisymplectic groupoid first. Then the Morita invariance principle guarantees that the resulting quantization does not depend on the particular choice of Morita-equivalent quasi-symplectic groupoid. As a special case, when is the AMM quasi-symplectic groupoid, our construction yields the prequantization of quasi-Hamiltonian G-spaces of Alekseev–Malkin–Meinrenken and their symplectic reductions, and our quantization condition coincides with that of Alekseev–Meinrenken [2]. Quantization of Hamiltonian spaces for symplectic groupoids was studied in [21]. Note that in the usual Hamiltonian case, since the symplectic 2-form defines a zero class in the third cohomology group of the groupoid T ∗ G ⇒ g∗ , which is the equivariant cohomology HG3 (g∗ ), gerbes do not appear explicitly. However, for a general quasi-symplectic groupoid (for instance the AMM quasi-symplectic groupoid), since the 3-cocycle ω + may define a nontrivial class, gerbes are inevitable in the construction. Also note that no nondegeneracy condition is needed in the quantization construction, so we drop this assumption in the present paper to assure full generality. This paper is organized as follows. In Section 2, we review some basic results concerning pre-quasi-symplectic groupoids and their Hamiltonian spaces. In Sec-

Quantization of pre-quasi-symplectic groupoids

425

tion 3, we gather some important results on S 1 -bundles and S 1 -central extensions. We give a simple formula for the index of an S 1 -bundle over a central extension in terms of the Chern class. In Section 4, we introduce prequantizations of pre-quasisymplectic groupoids and discuss compatible prequantizations of their Hamiltonian spaces. Section 5 is devoted to the description of a geometric integrality condition of pre-Hamiltonian -spaces. The application to quasi-Hamiltonian G-spaces is discussed. Unless specified, by a groupoid in this paper, we always mean a Lie groupoid whose orbit space is connected. A remark is in order concerning terminology. In [7], quasi-symplectic groupoids are called presymplectic groupoids, where some “nondegeneracy’’ condition is assumed. Here we choose to use the “quasi’’ part of the terminology to refer to the presence of a 3-form and to use “pre-’’ to mean that “nondegeneracy’’ is flexible. Note that it would be interesting to investigate what notion of polarization would be relevant for the next step of this quantization scheme. Prequantization of symplectic groupoids was first studied by Alan Weinstein and the second author in [19], when the second author was his Ph.D. student. In the same paper, S 1 -central extensions of Lie groupoids were also systematically investigated for the first time. Undoubtedly,Alan Weinstein’s work and insights have had a tremendous impact on the development of this subject in the past two decades. It is our great pleasure to dedicate this paper to him.

2 Pre-Hamiltonian -spaces and classical intertwiner spaces 2.1 Pre-quasi-symplectic groupoids and their pre-Hamiltonian spaces First, let us recall the definition of the de Rham double complex of a Lie groupoid. Let ⇒ M be a Lie groupoid. Define for all p ≥ 0 p = ×M · · · × M , :; < 9 p times

i.e., p is the manifold of composable sequences of p arrows in the groupoid ⇒ M (and 0 = M). We have p + 1 canonical maps p → p−1 (each leaving out one of the p + 1 objects involved in a sequence of composable arrows), giving rise to a diagram / / / 1 (1) · · · 2 / 0 . / • Consider the double complex (• ): · ·O ·

· ·O ·

d

1 ( O 0)

d ∂

d

0 (0 )

· ·O ·

/ 1 ( ) O 1

d ∂

d ∂

/ 0 ( ) 1

(2)

/ 1 ( ) O 2

∂

/ ···

∂

/ ···

d ∂

/ 0 ( ) 2

426


Its boundary maps are d : k (p ) → k+1 (p ), the usual exterior derivative of differentiable forms and ∂ : k (p ) → k (p+1 ), the alternating sum of the pullback maps of (1). We denote the total differential by δ = (−1)p d + ∂. The cohomology • groups of the total complex CdR (• ) k HdR (• ) = H k ( • (• ))

are called the de Rham cohomology groups of ⇒ M. Definition 2.1. A pre-quasi-symplectic groupoid is a Lie groupoid ⇒ M equipped with a 2-form ω ∈ 2 () and a 3-form ∈ 3 (M) such that d = 0,

dω = ∂ ,

and

∂ω = 0.

(3)

In other words, ω + is a 3-cocycle of the total de Rham complex of the groupoid ⇒ M. A pre-quasi-symplectic groupoid ( ⇒ M, ω + ) is said to be exact if is an exact 3-form on M. A quasi-symplectic groupoid is a pre-quasi-symplectic groupoid ( ⇒ M, ω +

), where ω satisfies a certain nondegenerate condition [7, 22]. Quasi-symplectic groupoids are natural generalization of symplectic groupoids, whose momentum map theory unifies various momentum map theories, including the ordinary Hamiltonian G-spaces, Lu’s momentum maps of Poisson group actions, and group-valued momentum maps of Alekseev–Malkin–Meinrenken. Definition 2.2. Given a pre-quasi-symplectic groupoid ( ⇒ M, ω + ), a preHamiltonian -space is a (left) -space J : X → M (i.e., acts on X from the left) with a compatible 2-form ωX ∈ 2 (X) such that (1) dωX = J ∗ ; (2) the graph of the action = {(r, x, rx)|t (r) = J (x)} ⊂ × X × X (where X is the manifold X endowed with the form −ωX ) is isotropic with respect to the 2-form (ω, ωX , −ωX ). To illustrate the intrinsic meaning of the above compatibility condition, let us elaborate it in terms of groupoids. Let ×M X ⇒ X be the transformation groupoid corresponding to the -action, and, by abuse of notation, J : ×M X → the natural projection. It is simple to see that ×M X X

J

/

J

/M

(4)

is a Lie groupoid homomorphism. Therefore, it induces a map, i.e., the pullback map, on the level of the de Rham complex: J ∗ : • (• ) → • (( ×M X)• ).


427

Proposition 2.3 ([22]). Let ( ⇒ M, ω + ) be a pre-quasi-symplectic groupoid and J : X → M a left -space. A 2-form ωX ∈ 2 (X) is compatible with the action if and only if J ∗ (ω + ) = δωX . (5) 2.2 Classical intertwiner spaces Consider a pre-quasi-symplectic groupoid ( ⇒ M, ω + ), and pre-Hamiltonian J1

J2

spaces (X1 → M, ω1 ), and (X2 → M, ω2 ). Assume that \(X2 ×M X1 ) is a smooth manifold, and denote by p : X2 ×M X1 → \(X2 ×M X1 ) the natural projection. Note that i ∗ (−ω2 , ω1 ), where i : X2 ×M X1 → X2 × X1 is the natural embedding, is a closed 2-form on X2 ×M X1 . Proposition 2.4. The 2-form i ∗ (−ω2 , ω1 ) descends to a closed 2-form on \(X2 ×M X1 ). Therefore, \(X2 ×M X1 ) is a presymplectic manifold. To prove this proposition, we need a technical lemma. Lemma 2.5 ([11]). Let ⇒ M be a Lie groupoid and X → M a left -space. Assume that \X is a smooth manifold. A differential form ω ∈ ∗ (X) descends to a differential form on the quotient \X if and only if ∂ω = 0, where ∂ is with respect to the transformation groupoid ×M X ⇒ X. Proof of Proposition 2.4. Note that the manifold X2 ×M X1 with the momentum map J : X2 ×M X1 → M, J (x2 , x1 ) = J1 (x1 ) = J2 (x2 ), is naturally a -space, where ⇒ M acts on X2 ×M X1 diagonally. Then ∂[i ∗ (−ω2 , ω1 )] = i ∗ (−∂ω2 , ∂ω1 ) = i ∗ (−J2∗ ω, J1∗ ω)

= ((J2 × J1 ) ◦ i)∗ (−ω, ω)

= 0, where J1 , J2 and i are, respectively, the groupoid homomorphisms: × M Xk Xk

Jk

Jk

/ k = 1, 2.

(6)

/M

and ×M (X1 ×M X2 ) X1 ×M X2

/ ( ×M X1 ) × ( ×M X2 ) ,

i

i

/ X1 × X 2

(7)

428


and ∂[i ∗ (−ω2 , ω1 )] and ∂ωk , k = 1, 2, are with respect to the groupoids on the left-hand side of equations (7) and (6), respectively. The conclusion thus follows from Lemma 2.5.

The presymplectic manifold \(X2 ×M X1 ) is called the classical intertwiner space and is denoted by X2 × X1 for simplicity. In particular, if ( ⇒ M, ω + ) is J1

J2

a quasi-symplectic groupoid and (X1 → M, ω1 ) and (X2 → M, ω2 ) are Hamiltonian -spaces, and if J1 : X1 → M and J2 : X2 → M are clean, then X2 × X1 becomes a symplectic manifold. See [22] for details.

3 S 1 -bundles and S 1 -central extensions In this section we recall some basic results concerning S 1 -bundles and S 1 -central extensions over a Lie groupoid. For details, consult [4, 5, 18]. 3.1 Integral de Rham cocycles Let us recall some basic facts concerning singular homology. For any manifold N , we denote by (C• (N, Z), d) the piecewise smooth singular chain complex, and Zk (N, Z) the space of smooth k-cycles. For a smooth map φ : M → N , we denote by φ∗ both the chain map from (C• (M, Z), d) to (C• (N, Z), d) and the morphism of singular homology H∗ (M, Z) → H∗ (N, Z) induced by φ. For any Lie groupoid ⇒ 0 , consider the double complex C• (• , Z): ··· ↓d

··· ↓d

··· ↓d

∂

∂

∂

∂

C1 (0 , Z) ← C1 (1 , Z) ← C1 (2 , Z) ↓d ↓d ↓d C0 (0 , Z) ← C0 (1 , Z) ← C0 (2 , Z), where 0 = M, and ∂ : Ck (p , Z) → Ck (p−1 , Z) is the alternating sum of the chain maps induced by the face maps. We denote the total differential by δ = (−1)p d + ∂. Its homology will be denoted by Hk (• , Z). By Zk (• , Z) we denote the space of k-cycles and by [C] ∈ H∗ (• , Z) the class of a given cycle C. Note that Ck (p , Z) is the free Abelian group generated by the piecewise smooth maps k → p . The construction above can be carried out in exactly the same way replacing Z by R. The corresponding homology groups are denoted by Hk (• , R). According to the universal-coefficient formula (see, for example, [17]), there is a canonical isomorphism Hk (• , R) ! Hk (• , Z) ⊗Z R. • There is a natural pairing between C• (• , R) and CdR (• ) given as follows. For any generator C : k → p in C• (• , Z), + C ∗ ω if ω ∈ k (p ), k C, ω = (8) 0 otherwise.


429

For simplicity, we will denote this pairing by C ω. With this notation, the pairing satisfies the following identities: ω = dω, dC

C

ω= ∂C

C

ω= δC

(9)

∂ω,

δω. C

Moreover, if φ : G → H is a groupoid homomorphism, then for any C ∈ • C• (G• , R) and ω ∈ CdR (H• ), ω = φ ∗ ω. (10) φ∗ (C)

C

The following result is standard (see, for example, [8, Proposition 6.1]). k ( ) → R, ([C], [ω]) → Proposition 3.1. The pairing Hk (• , R) ⊗ HdR • nondegenerate.

Let k ZdR (• , Z)

C

ω is

= {ω ∈

k ZdR (• )

|

ω ∈ Z for any cycle C ∈ Zk (• , Z)}.

(11)

C k ( , Z) are called integral de Rham cocycles, or simply integral Elements in ZdR • cocycles.

3.2 S 1 -bundles and S 1 -central extensions In this subsection, we recall some basic notations and results concerning S 1 -bundles and S 1 -central extensions over a Lie groupoid. For details, see [4, 5]. Definition 3.2. Let ⇒ M be a Lie groupoid. A (right) S 1 -bundle over ⇒ M is a (right) S 1 -bundle P over M, together with a (left) action of on P which respects the S 1 -action (i.e., we have (γ · x) · t = γ · (x · t) for all t ∈ S 1 and all compatible pairs (γ , x) ∈ ×M P ). Let Q ⇒ P denote the corresponding transformation groupoid ×M P ⇒ P . There is a natural groupoid homomorphism π from Q ⇒ P to ⇒ M. Of course, Q is an S 1 -bundle over . 1 (Q ), where θ ∈ 1 (P ) is a conA pseudo-connection is a 1-cochain θ ∈ CdR • 2 (Q ) descends to nection 1-form for the S 1 -bundle P → M. One checks that δθ ∈ CdR •

430


2 ( ). In other words, there exist unique ω ∈ 1 () and ∈ 2 (M) a 2-cocycle in ZdR • such that δθ = π ∗ (ω + ).

Then ω + is called the pseudo-curvature, which is an integral 2-cocycle. Its class [ω + ] ∈ H 2 (• , Z) is called the Chern class of the S 1 -bundle P . Proposition 3.3 ([4, 5]). Let ⇒ M be a proper Lie groupoid. Assume that ω + ∈ 2 ( ) is an integral 2-cocycle. Then there exists an S 1 -bundle

1 () ⊕ 2 (M) ⊂ CdR • P over ⇒ M and a pseudo-connection θ ∈ 1 (P ) for the bundle P → M whose pseudo-curvature equals ω + . Definition 3.4. Let ⇒ M be a Lie groupoid. An S 1 -central extension of ⇒ M consists of (1) a Lie groupoid R ⇒ M, together with a morphism of Lie groupoids (π, id) : [R ⇒ M] → [ ⇒ M], (2) a left S 1 -action on R, making π : R → a (left) principal S 1 -bundle. These two structures are compatible in the sense that (s · x)(t · y) = st · (xy) for all s, t ∈ S 1 and (x, y) ∈ R ×M R. Given an S 1 -central extension R of ⇒ M, a pseudo-connection is a 2-cochain 2 (R ), where θ ∈ 1 (R) is a connection 1-form for the bundle R → θ + B ∈ CdR • and B ∈ 2 (M). It is simple to check that δ(θ + B) descends to a 3-cocycle in Z 3 (• ), i.e., δ(θ + B) = π ∗ (η + ω + ) 3 ( , Z) for some η + ω + ∈ Z 3 (• ). Then η + ω + is an integral cocycle in ZdR • 3 and it is called the pseudo-curvature. Its class [η + ω + ] ∈ H (• , Z) is called the Dixmier–Douady class of R.

Proposition 3.5 ([4, 5]). Assume that ⇒ M is a proper Lie groupoid. Given any 3 ( ) such that 3-cocycle η + ω + ∈ ZdR • (1) [η + ω + ] is integral, and (2) is exact, there exists a Lie groupoid S 1 -central extension R ⇒ M of the groupoid ⇒ M and a pseudo-connection θ + B ∈ 1 (R) ⊕ 2 (M) such that its pseudo-curvature equals η + ω + . 3.3 Index of an S 1 -bundle over a central extension π

p

Let R → ⇒ M be an S 1 -central extension, and S 1 → L → M a principal S 1 bundle over the groupoid R ⇒ M with Chern class [L] ∈ H 1 (R• , S 1 ). The example below will be useful in the future. Example 3.6. Consider, for any k ∈ Z, the principal S 1 -bundle Bk : S 1 → · over S 1 ⇒ ·, where the groupoid S 1 ⇒ · acts on Bk by


λ · z = λk z

∀λ ∈ S 1 ⇒ · and

431

∀z ∈ S 1 → ·.

It is well known that H 1 (S•1 , S 1 ) ! Z. Under this isomorphism, the class [Bk ] is simply equal to k. It is also simple to see that the Chern class of Bk can be represented by k where

dt 2π

dt ∈ Z 1 (S 1 ) ⊂ Z 2 ((S 1 )• ), 2π

(12)

is the normalized Haar measure on S 1 .

For any m ∈ M, there exists a groupoid homomorphism fm from S 1 ⇒ · to R ⇒ M defined by fm (λ) = λ · 1m ∀λ ∈ S 1 , (13) where 1m ∈ R is the unit element over m ∈ M. This homomorphism induces a map fm∗ : H 1 (R• , S 1 ) → H 1 (S•1 , S 1 ) ! Z.

(14)

For a principal S 1 -bundle L over R ⇒ M, we define its index by Ind m (L) = fm∗ ([L]) ∈ H 1 (S•1 , S 1 ) ! Z. We list some of its important properties below. p

π

Proposition 3.7. Let R → ⇒ M be an S 1 -central extension, and S 1 → L → M an (right) principal S 1 -bundle over the groupoid R ⇒ M. Then (1) the index is characterized by the relation fm (λ) · l = l · λIndm (L) ∀λ ∈ S 1 ,

l ∈ p −1 (m),

where the dot on the left-hand side denotes the R-action on L, while the dot on the right-hand side refers to the S 1 -action on L; (2) for any m ∈ M, the pullback fm∗ L is isomorphic to BIndm (L) ; (3) Ind m (L) is constant on the groupoid orbits; (4) Ind m (L) is constant on any connected component of M; and (5) if \M is path connected, then the index Ind m (L) is independent of m ∈ M. Proof. (1), (2) Let l be any point in the fiber Lm = p −1 (m). For any λ ∈ S 1 , there exists a unique φ(λ) ∈ S 1 such that fm (λ) · l = l · φ(λ).

(15)

The map λ → φ(λ) does not depend on the choice of l in the fiber p−1 (m) and is a group homomorphism from S 1 to S 1 . Therefore, it is of the form φ(λ) = λk for some k ∈ Z.

432


Now fm∗ ([L]) ∈ H 1 (S•1 , S 1 ) is the Chern class associated to the pullback of L by fm . On the other hand, according to equation (15), fm∗ L is isomorphic (as a principal S 1 -bundle over S 1 ⇒ ·) to Bk . Therefore, k = Ind m (L) and equation (15) implies fm (λ) · l = l · λIndm (L)

∀l ∈ p−1 (m).

(16)

This proves (1) and (2). (3) For any γ ∈ R with s(γ ) = n and t (γ ) = m, we have γ 1m = 1n γ . It follows from equation (13) that γfm (λ) = fn (λ)γ . Now for any l ∈ p −1 (m), we have (γfm (λ)) · l = (fn (λ)γ ) · l. On one hand, we have (γfm (λ)) · l = (γ · l) · λIndm (L) ,

(17)

(fn (λ)γ ) · l = fn (λ)(γ · l) = (γ · l) · λIndn (L) .

(18)

and From equations (17) and (18), it follows that Ind m (L) = Ind n (L). (4) It is clear from equations (16) that Ind m (L) depends continuously on m ∈ M. Since it is a Z-valued function, we have Ind m (L) = Ind n (L) for any pair of points (m, n) ∈ M × M that are in the same connected component of M. (5) This follows from (3) and (4) immediately.

3.4 Index and Chern class From now on, we will assume that the space of orbits M/ is path-connected, and denote the index of L simply by Ind(L). Therefore, we have a group homomorphism: Ind(L) : H 1 (R• , S 1 ) → Z. From the commutativity of the diagram i

H 1 (R• , S 1 ) → H 2 (R• , Z) ↓ ↓ , i

H 1 (S•1 , S 1 ) → H 2 (S•1 , Z) we see that Ind(L) factors through H 2 (R• , Z) → Z. In the following proposition, we give an explicit formula for Ind(L) in terms of the Chern class. Proposition 3.8. Assume that L → M is a principal S 1 -bundle over R ⇒ M with the π 2 (R , Z), where R → Chern class [θ + ω] ∈ HdR ⇒ M is an S 1 -central extension, • 1 2 and θ + ω ∈ (R) ⊕ (M). Then the index of L is given by Ind(L) = θ, π −1 ((m))

where : M → is the unit map.


433

Proof. Let L be the pullback of the principal S 1 -bundle L via the homomorphism fm : S 1 → R. The Chern class of L is the pullback of the Chern class of L, i.e., 2 (S 1 ). Since f ∗ ω is a 2-form over a point, it the class defined by fm∗ θ + fm∗ ω ∈ CdR • m vanishes and therefore the Chern class of L is represented by fm∗ θ ∈ 1 (S 1 ). By Proposition 3.7, L is isomorphic to BInd(L) . According to equation (12), the dt dt identity fm∗ θ = Ind(L) 2π + δg = Ind(L) 2π + dg holds for some function g ∈ C ∞ (S 1 , R). Now since fm is a bijection from S 1 to π −1 ((m)), we have θ = fm∗ θ. π −1 ((m))

Therefore,

θ=

π −1 ((m))

fm∗ θ

S1

= Ind(L)

S1

S1

dt + 2π

dg = Ind(L).

S1

Recall that a line bundle L → M over R ⇒ M is called a (, R)-twisted line bundle if Ker π ∼ = M × S 1 acts on L by scalar multiplication, where S 1 is identified with the unit circle in C [18]. The following corollary is an immediate consequence of Proposition 3.8 and Proposition 3.7. Corollary 3.9. Under the hypotheses of Proposition 3.8, the S 1 -bundle L → M defines a (, R)-twisted line bundle if and only if θ = 1. π −1 ((m))

4 Prequantization of classical intertwiner spaces 4.1 Compatible prequantizations Definition 4.1. A prequantization of a pre-quasi-symplectic groupoid ( ⇒ M, ω + π

) consists of an S 1 -central extension R → ⇒ M together with a pseudoconnection θ + B ∈ 1 (R) ⊕ 2 (M) such that δ(θ + B) = π ∗ (ω + ).

(19)

According to Proposition 3.3, if ⇒ M is a proper Lie groupoid, a prequantization exists if and only if ( ⇒ M, ω + ) is exact and ω + is an integral 3-cocycle. A pre-quasi-symplectic groupoid ( ⇒ M, ω + ) is said to be integral if ω + is an integral cocycle. Definition 4.2. Let ( ⇒ M, ω + ) be an exact pre-quasi-symplectic groupoid and J

(R → ⇒ M, θ + B) a prequantization. Assume that (X → M, ωX ) is a preHamiltonian -space. A compatible prequantization of X consists of an S 1 -bundle φ : L → X with a connection 1-form θL ∈ 1 (L) such that

434


(1) J˜ = J ◦ φ : L −→ M is a left R-space and the action satisfies (s · κ)(t · x) = st · (κx) for all s, t ∈ S 1 and (κ, x) ∈ R ×M X a compatible pair; (2) the 1-form (θ, θL , −θL ) ∈ 1 (R × L × L) vanishes on the graph of the action + = {(κ, l, κl)|κ ∈ R, l ∈ L compatible pairs}; and (3) dθL = φ ∗ (J ∗ B − ωX ). Note that the second condition above is equivalent to saying that (R × L × p L)/T 2 −→ × X × X with p([κ, l, m]) = (π(κ), φ(l), φ(m)) is a flat S 1 -bundle ¯ which is the 1-form on (R × L × L)/T 2 naturally induced with the connection ', from ' = (θ, θL , −θL ) ∈ 1 (R × L × L) (see [21]). Example 4.3. If is the symplectic groupoid (T ∗ G ⇒ g∗ , ω), where ω ∈ 2 (T ∗ G) is the canonical cotangent symplectic 2-form, a prequantization of can be taken to be R ∼ = T ∗ G × S 1 → T ∗ G, the trivial S 1 -bundle and θ = θT ∗ G + dt, where ∗ θT G ∈ 1 (T ∗ G) is the Liouville 1-form and t is the natural coordinate on S 1 . A Hamiltonian -space is a Hamiltonian G-space J : X → g∗ in the usual sense. It is simple to see that a compatible pre-quantization is a G-equivariant prequantization of X, which always exists when G is connected and simply connected [10]. More generally, the following result was proved in [21]. (The theorem was stated for the symplectic case, but it is valid for the presymplectic case as well.) Proposition 4.4. Let ( ⇒ M, ω) be an s-connected and s-simply connected preJ

symplectic groupoid and (X → M, ωX ) a pre-Hamiltonian space. If both ω and ωX 2 () and H 2 (X), respectively, then represent integral cohomology classes in HdR dR there exists a compatible prequantization. For a given pre-quasi-symplectic groupoid ( ⇒ M, ω+ ) and a prequantization (R → ⇒ M, θ +B), let ×M X ⇒ X be the transformation groupoid as in equation (4). By pulling back the S 1 -central extension R → ⇒ M via J , one obtains an S 1 -central extension of groupoids R ×M X → ×M X ⇒ X. Here R ×M X is again a transformation groupoid, where R acts on X by projecting R to and using the given -action on X. By abuse of notation, we still use J to denote the projection R ×M X → R. Therefore, we have the following homomorphism of S 1 -central extensions of groupoids: J

/R

×M X

J

/

X

J

/M

R ×M X

(20)


435

Remark 4.5. Note that Proposition 2.3 implies that the Dixmier–Douady class of R ×M X → ×M X ⇒ X vanishes. If ⇒ M is a proper groupoid, so is ×M X ⇒ X. Therefore, R ×M X → ×M X ⇒ X defines a trivial S 1 -gerbe. According to Proposition 4.2 of [4], there exists an S 1 -bundle E → X such that R ×M X ∼ = s ∗ E ⊗ t ∗ E as a central extension. Proposition 4.6. Let ( ⇒ M, ω + ) be an exact pre-quasi-symplectic groupoid J

and (R → ⇒ M, θ + B) its prequantization. Assume that (X → M, ωX ) is a φ

pre-Hamiltonian -space. Then (L → X, θL ) is a compatible prequantization of X if and only if (the associated line bundle of ) φ : L → X is a twisted line bundle over R ×M X → ×M X ⇒ X with the pseudo-connection and the pseudo-curvature being given by θL and J ∗ θ + (J ∗ B − ωX ) ∈ 1 (R ×M X) ⊕ 2 (X), respectively. φ

Proof. Given a compatible prequantization L → X, define an action of R×M X ⇒ X on L by (κ, φ(l)) · l = κl, where κ ∈ R and l ∈ L are compatible pairs. It is simple to φ

check that all the compatibility conditions are satisfied so that L → X is a twisted line bundle over the S 1 -central extension R ×M X → ×M X ⇒ X. It is simple to see that the corresponding transformation groupoid (R ×M X) ×X L ⇒ L is isomorphic to the transformation groupoid R ×M L ⇒ L. Moreover, it is simple to see that Condition (2) of Definition 4.2 implies that ∂θL = φ ∗ J ∗ θ,

(21)

where, by abuse of notation, we use φ to denote the Lie groupoid homomorphism: R ×M L L

φ

/ R ×M X

(22)

/X

φ

and ∂θL is with respect to the groupoid R ×M L ⇒ L. Therefore, we have δθL = ∂θL + dθL = φ ∗ (J ∗ θ + J ∗ B − ωX ). The converse can be proved by working backwards.

As an immediate consequence, we have the following. Corollary 4.7. Under the hypotheses of Proposition 4.6 and assuming that ⇒ M is J

proper, for a pre-Hamiltonian -space (X → M, ωX ), a compatible prequantization 2 ((R × X) , Z). exists if and only if J ∗ (θ + B) − ωX is an integral 2-cocycle in ZdR M • Proof. One direction is obvious by Proposition 4.6. For the other direction, note that Proposition 2.3 implies that J ∗ (θ + B) − ωX is always a 2-cocycle since δ(J ∗ (θ + B) − ωX ) = J ∗ δ(θ + B) − π ∗ δωX = J ∗ π ∗ (ω + ) − π ∗ J ∗ (ω + ) = 0.

436


Here we have used equations (19) and (6). If J ∗ (θ + B) − ωX is an integral cocycle in 2 ((R × X) , Z), according to Proposition 3.3, there exists an S 1 -bundle L → X ZdR M • over R ⇒ X and a pseudo-connection θL ∈ 1 (L) whose pseudo-curvature equals to J ∗ θ + (J ∗ B − ωX ). According to Corollary 3.9, one sees that (the associated line bundle of) L is indeed a twisted line bundle over R ×M X → ×M X ⇒ X. Then L → X is a compatible prequantization by Proposition 4.6.

4.2 Prequantization of classical intertwiner spaces We are now ready to state the main theorem of this section. Theorem 4.8. Let ( ⇒ M, ω + ) be an exact pre-quasi-symplectic groupoid Jk

and (R → ⇒ M, θ + B) a prequantization. Assume that (Xk → M, ωk ), k = 1, 2, are pre-Hamiltonian -spaces, ⇒ M acts freely on X2 ×M X1 and φk

X2 × X1 = \(X2 ×M X1 ) is a smooth manifold. Let (Lk → Xk , θk ), be a compatible prequantization of Xk for k = 1, 2. Then φ : R\(L2 ×M L1 ) → X2 × X1 ,

φ[l2 , l1 ] = [φ2 (l2 ), φ1 (l1 )],

with the S 1 -action λ · [l2 , l1 ] = [λ · l2 , l1 ], λ ∈ S 1 , is an S 1 -principal bundle. Moreover, i ∗ (θ2 , −θ1 ) descends to a connection 1-form on R\(L2 ×M L1 ), which defines a prequantization of the classical intertwiner space X2 × X1 . Here i : L2 ×M L1 → L2 × L1 is the natural embedding. Proof. One checks directly that φ : R\(L2 ×M L1 ) → X2 × X1 is an S 1 -bundle. Now let R ⇒ M act on L2 ×M L1 diagonally. We have ∂i ∗ (θ2 , −θ1 ) = i ∗ (∂θ2 , −∂θ1 ) = i ∗ (φ2∗ J2∗ θ, −φ1∗ J1∗ θ ) = 0. Hence i ∗ (θ2 , −θ1 ) descends to a 1-form on the quotient space R\(L2 ×M L1 ), which can be easily seen to be a connection 1-form. Now d(i ∗ (θ2 , −θ1 )) = i ∗ (dθ2 , −dθ1 ) = i ∗ (φ2∗ (J2∗ B − ω2 ), φ1∗ (J1∗ B − ω1 )) = i ∗ (φ2 × φ1 )∗ (−ω2 , ω1 ),

where in the last equality we used the relation J1 ◦ φ1 = J2 ◦ φ2 on L2 ×M L1 . Here φk and Jk , k = 1, 2 are groupoid homomorphisms: R ×M Lk Lk

φk

φk

and i is the groupoid homomorphism:

/ R × M Xk / Xk

Jk

/R

Jk

/M

(23)


R ×M (L2 ×M L1 ) L2 × M L1

i

/ (R ×M L2 ) × (R ×M L1 )

i

/ L2 × L 1

437

(24)

This completes the proof. 4.3 Morita equivalence

Definition 4.9. Pre-quasi-symplectic groupoids (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) are said to be Morita equivalent if there exists a Morita equivalence ρ σ bimodule G0 ← X → H0 between the Lie groupoids G and H , together with a ρ×σ

2-form ωX ∈ 2 (X) such that (X → G0 × H0 , ωX ) is a pre-Hamiltonian G × H space, where the G×H -action on X is given by (g, h)·x = gxh−1 for all compatible triples g ∈ G, h ∈ H , and x ∈ X. One easily checks that this is indeed an equivalence relation among pre-quasisymplectic groupoids. Let Q ⇒ X be the transformation groupoid Q : (G × H ) ×(G0 ×H0 ) X ⇒ X. Then the natural projections pr 1 : Q → G and pr 2 : Q → H are groupoid homomorphisms. As an immediate consequence of Proposition 2.3, we have the following identity pr ∗1 (ωG + G ) − pr ∗2 (ωH + H ) = δωX . Note that the axioms of Morita equivalence of Lie groupoids assure that, as groupoids, Q∼ = G[X] and Q ∼ = H [X] (see the proof of [22, Proposition 4.5]), where G[X] ⇒ X and H [X] ⇒ X are the pullback groupoids of G and H using ρ and σ , respectively. Recall that for a given Lie groupoid ⇒ M, two cohomologous 3-cocycles ωi + i ∈ 2 () ⊕ 3 (M), i = 1, 2, are said to differ by a gauge transformation of the first type if (ω1 + 1 ) − (ω2 + 2 ) = δB for some B ∈ 2 (M). By a Morita morphism from the pre-quasi-symplectic groupoid ( ⇒ M , ω +

) to ( ⇒ M, ω+ ), we mean a Morita morphism of the Lie groupoid p : → (i.e., is isomorphic to the pullback groupoid [M ] ⇒ M ) such that ω + and p∗ ω + p ∗ differ by a gauge transformation of the first type. The following result gives a more intuitive explanation of Morita equivalence. Proposition 4.10. Two pre-quasi-symplectic groupoids are Morita equivalent if and only if there exists a third pre-quasi-symplectic groupoid together with a Morita morphism to each of them.

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Corollary 4.11. For two Morita-equivalent pre-quasi-symplectic groupoids, if one is integral, so is the other. Therefore, Morita equivalence induces an equivalence relation among integral pre-quasi-symplectic groupoids. One of the most important features of Morita-equivalent pre-quasi-symplectic groupoids is the following. Theorem 4.12. Suppose that (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) are Morita-equivalent pre-quasi-symplectic groupoids with an equivalence bimodule ρ σ G0 ← X → H0 . Then we have the following: (1) Corresponding to any pre-Hamiltonian G-space JF : F → G0 , there is a unique (up to isomorphism) pre-Hamiltonian H -space JE : E → H0 such that F and E are a pair of related pre-Hamiltonian spaces and vice versa. (2) Let JFi : Fi → G0 , i = 1, 2, be pre-Hamiltonian G-spaces and JEi : Ei → H0 , i = 1, 2, their related pre-Hamiltonian H -spaces. Then F2 ×G F1 and E2 ×H E1 are diffeomorphic as presymplectic manifolds (in the sense that if one is smooth so is the other). Proof. This was proved in [22] for quasi-symplectic groupoids and their Hamiltonian spaces. One can prove this theorem in a similar fashion (in fact in a simpler way by using Proposition 2.4). We will leave the details to the reader.

We now can introduce Morita equivalence for the prequantization of pre-quasisymplectic groupoids. Definition 4.13. Let (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) be Moritaequivalent integral exact pre-quasi-symplectic groupoids with an equivalence bimodρ σ ule (G0 ← X → H0 , ωX ). We say their prequantizations (RG → G ⇒ G0 , θG +BG ) and (RH → H ⇒ H0 , θH + BH ) are Morita equivalent if X admits a compatible prequantization (Z → X, θZ ) with respect to the prequantization of the pre-quasisymplectic groupoid (RG ×RH )/S 1 → G×H ⇒ G0 ×H0 , (θG +θH )+(BG +BH )). It is simple to see that G0 ←Z→H0 is an equivalence bimodule of S 1 -central extensions in the sense of [18, Definition 2.11]. Remark 4.14. 1. Note that prequantizations can be Morita equivalent as S 1 -central extensions, but not Morita equivalent as prequantizations. The former simply means that they correspond to isomorphic S 1 -gerbes, and up to a torsion, are determined by their Dixmier–Douady classes. 2. It would be interesting to investigate the following question: given two Moritaequivalent pre-quasi-symplectic groupoids and a prequantization of one of them, is it possible to construct a Morita-equivalent prequantization for the other prequasi-symplectic groupoid?


439

A useful feature of Morita equivalence is that it gives a recipe which allows us to construct compatible prequantizations. Theorem 4.15. For Morita-equivalent prequantizations of pre-quasi-symplectic groupoids, there is an equivalence of categories of compatible prequantizations of pre-Hamiltonian spaces. Proof. Let (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) be Morita-equivalent ρ integral exact pre-quasi-symplectic groupoids with an equivalence bimodule (G0 ← σ X → H0 , ωX ), and (RG → G ⇒ G0 , θG + BG ) and (RH → H ⇒ H0 , θH + BH ) Morita-equivalent prequantizations given by (Z → X, θZ ).Assume that J : F → G0 is a pre-Hamiltonian G-space and (L → F, θL ) a compatible prequantization. It is J

known that the corresponding pre-Hamiltonian H -space is E := X ×G F → H0 , where J : E → H0 and the H -action on E are defined by J ([x, f ]) = σ (x) and h · [x, f ] = [x · h−1 , f ], respectively. Let L = Z ×RG L. Then it is clear that L is an S 1 -bundle over E, and RH acts on L equivariantly. It is simple to check that i ∗ (θZ , −θL ), where i : Z ×G0 L → Z × L, descends to a 1-form on the quotient space Z ×RG L, which is indeed a connection 1-form θL on L . It is routine to check that (L → E, θL ) is a compatible prequantization of the pre-Hamiltonian H -space J : E → H0 . The inverse functor can be constructed in a similar fashion.

Remark 4.16. The above theorem indicates a useful method which enables one to transform prequantizations of Hamiltonian LG-spaces to prequantizations of quasiHamiltonian G-spaces of AMM and vice versa. The latter is understood as a compatible prequantization corresponding to the quasi-symplectic groupoid (G × G)[U] ⇒ H Ui , which is the pullback quasi-symplectic groupoid of the AMM quasi-symplectic groupoid using an open covering U = (Ui )i∈I of G (seeH[14], for instance, for an explicit construction). It is known that (G × G)[U] ⇒ Ui is Morita equivalent to the symplectic groupoid (LG × Lg ⇒ Lg, ωLG×Lg ) according to Proposition 4.26 [22]. The question is therefore boiled down to the construction of a compatible prequantization of the Morita equivalence Hamiltonian bimodule.

5 Integral pre-Hamiltonian -spaces The main purpose of this section is to give a geometric integrality condition which guarantees the existence of a prequantization of a pre-Hamiltonian -space. 5.1 Integrality condition Lemma 5.1. Let J : G → H be a groupoid homomorphism. By Ker(J∗ ), we de2 (G ). The following note the kernel of J∗ : H2 (G• , Z) → H2 (H• , Z). Let ω ∈ ZdR • conditions are equivalent: 2 (H ) such that (1) There exists + ∈ ZdR •

440

C. Laurent-Gengoux and P. Xu 2 ω + J ∗ + ∈ ZdR (G• , Z).

(2) For any C ∈ Z2 (G• , Z) with [C] ∈ Ker(J∗ ), we have ω ∈ Z. C

Proof. (1) ⇒ (2): By definition, we have for any C ∈ Z2 (G• , Z), (ω + J ∗ +) ∈ Z.

(25)

C

From equation (9), we also have ∗ (ω + J +) = ω + C

C

+.

J∗ (C)

If [J∗ (C)] = 0, i.e., J∗ (C) = δD for some D ∈ C3 (H• , Z), then ∗ (ω + J +) = ω + + = ω + δ+ = ω C

C

δD

C

D

C

since δ+ = 0. Therefore, C ω ∈ Z. (2) ⇒ (1): Since there exists a Z-submodule H in H2 (G• , Z) such that H2 (G• , Z) = H ⊕ Ker(J∗ ), the Z-map f : Ker(J∗ ) → Z, f ([C]) = ω ∀[C] ∈ Ker(J∗ ), C

can be extended to a Z-map f˜ : H2 (G• , Z) → Z. According to Proposition 3.1, there 2 (G ) such that exists ω ∈ ZdR • f˜([C]) = ω ∀[C] ∈ H2 (G• , Z). C 2 (G , Z). Moreover, we have By equation (11), ω is an integral cocycle in ZdR • (ω − ω) = 0 ∀C ∈ Z2 (G• , Z) such that [C] ∈ Ker(J∗ ). (26) C 2 (H ) → H 2 (G ), we have Since J∗ : H2 (G• , R) → H2 (H• , R) is dual to J ∗ : HdR • • dR 2 ( ). This ⊥ ∗ ∗ Ker(J∗ ) = Im(J ). Therefore, [ω − ω] = J [+] for some + ∈ ZdR • proves (1).


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Definition 5.2. Let ( ⇒ M, ω + ) be a pre-quasi-symplectic groupoid. A preHamiltonian -space (X → M, ωX ) is said to satisfy the integrality condition if for any C ∈ Z2 (( ×M X)• , Z) and any D ∈ C3 (• , Z), δD = J∗ (C) ⇒ ωX − (ω + ) ∈ Z. (27) C

D

In this case, we also say that the pair (ωX , ω + ) satisfies the integrality condition. Remarks 5.3.

1. By taking C = 0, equation (27) implies that D (ω + ) ∈ Z ∀D ∈ Z3 (• , Z). That is, ω + must be an integral 3-cocycle and therefore ( ⇒ M, ω + ) must be an integral pre-quasi-symplectic groupoid. 2. If ω + is a 3-coboundary δK, then the integrality condition is equivalent to (ωX − J ∗ K) ∈ Z ∀C ∈ Z2 (( ×M X)• , Z) such that J∗ [C] = 0. (28) C

From now on, we shall always assume that ( ⇒ M, ω + ) is an integral pre-quasi-symplectic groupoid. The following lemma indicates that it is sufficient to require that equation (27) holds for a single representative (C, D) in every class of Ker(J∗ ). Lemma 5.4. Let ( ⇒ M, ω + ) be an integral pre-quasi-symplectic groupoid. A pre-Hamiltonian -space (X → M, ωX ) satisfies the integrality condition if and only if for any class c ∈ Ker J∗ , there exists C ∈ Z2 (( ×M X)• , Z) and D ∈ C3 (• , Z) with c = [C] and J∗ (C) = δD such that ωX − (ω + ) ∈ Z. C

D

Proof. Let C ∈ Z2 (( ×M X)• , Z) and D ∈ C3 (• , Z) be any pair satisfying J∗ (C ) = δD . Then [C ] ∈ Ker(J∗ ). By assumption, there exists a pair (C, D) such that [C] = [C ], J∗ (C) = δD, and C ωX − D (ω + ) ∈ Z. Assume that C = C + δE for some E ∈ C3 (( ×M X)• , Z). Then we have ⎛ ⎞ ωX − (ω + ) − ⎝ ωX − (ω + )⎠ C

D

=−

ωX +

δE

=−

C

(ω + ) − D

δωX + E

D

(ω + ) D

(ω + ) − D

(ω + ) D

442


J ∗ (ω + ) +

=− E

(ω + ) − D

D

=

(ω + )

(ω + ). D−J∗

(E)−D

Since δ(D − J∗(E) − D ) = J∗ (C − C − δE) = 0 and ω + is an integral cocycle,

it follows that D−J∗ (E)−D (ω + ) ∈ Z. This completes the proof. Now assume that ( ⇒ M, ω + ) is an integral exact pre-quasi-symplectic groupoid, and R → ⇒ M is a prequantization. Let θ + B ∈ 1 (R) ⊕ 2 (M) be a pseudo-connection satisfying equation (19). In order to fix the notation, recall that we have the following commutative diagram of groupoid homomorphisms J

R ×M X → R ↓π ↓π

(29)

J

×M X → where the horizontal arrows are projections. Lemma 5.5. Assume that C ∈ Z2 ((R ×M X)• , Z) satisfies J∗ (C ) = kZ + δD for some D ∈ C3 (R• , Z). Let C = π∗ (C ) and D = π∗ (D ). Then ωX − (ω + ) = k + (ωX − J ∗ (θ + B)), (30) C

C

D

where Z ∈ Z1 (R• , Z) is the 1-cycle defined by equation (42). Proof. First, since π : R ×M X → ×M X reduces to the identity map when being restricted to the unit spaces, we have ωX = ω X = ωX . (31) C

π∗ (C )

C

Now by equation (9), we have J ∗ (θ + B) = (θ + B) = k (θ + B) + (θ + B). C

J∗ (C )

Z

δD

According to Lemma 6.1, Z (θ + B) = Z θ = 1. Therefore, J ∗ (θ + B) = k + (θ + B) C

δD

=k+

δ(θ + B) (by equation (19)) D

(32)


=k+

π ∗ (ω + )

443

(by equation (9))

D

=k+

(ω + ). D

Hence it follows that ωX − (ω + ) = k + (ωX − J ∗ (θ + )). C

C

D

The following proposition gives a useful characterization of integrality condition. Proposition 5.6. Let ( ⇒ M, ω + ) be an integral pre-quasi-symplectic groupoid, J

and (R → ⇒ M, θ + B) a prequantization. Assume that (X → M, ωX ) is a preHamiltonian -space. Then the following conditions are equivalent: 2 ( ) such that (1) There exists a 2-cocycle + ∈ ZdR • 2 ((R ×M X)• , Z). ωX − J ∗ (θ + B) − J ∗ π ∗ + ∈ ZdR

(2) For any cycle C ∈ Z2 ((R ×M X)• , Z) such that [C ] ∈ Ker(π∗ ◦ J∗ ), we have (ωX − J ∗ (θ + B)) ∈ Z. C

(3) The pair (ωX , ω + ) satisfies the integrality condition. Proof. (1) ⇐⇒ (2): follows from Lemma 5.1. (2) ⇒ (3): Any class in Ker J∗ ⊂ H 2 (( ×M X)• , Z) can be represented by a 2-cocycle of the form C = π∗ (C ), where C ∈ Z2 ((R ×M X)• , Z). Then [C ] is in the kernel of J∗ ◦ π∗ = π∗ ◦ J∗ . It thus follows that [J∗ (C )] ∈ Ker(π∗ ). By Lemma 6.1, [J∗ (C )] = k[Z] for some k ∈ Z, where Z ∈ C1 (R• , Z) is defined by equation (42). In other words, there exists D ∈ C3 (R• , Z) such that J∗ (C ) = kZ + δD . Let D = π∗ (D ). One can easily see that δD = π∗ (J∗ (C )) = J∗ (C). Then by Lemma 5.5, we have C ωX − D (ω + ) ∈ Z. By Lemma 5.4, this implies that the pair (ωX , ω + ) satisfies the integrality condition. (3) ⇒ (2): Let C ∈ Z2 ((R × X)• , Z) be any cycle whose class is in the kernel of π∗ ◦ J∗ . Since [J∗ (C )] ∈ Ker(π∗ ), Lemma 6.1 implies that there exists k ∈ Z and D ∈ C3 (R• , Z) such that J∗ (C ) = kZ + δD . (33) Therefore, by equation (30), we have C (ωX −J ∗ (θ +B)) = −k+ C ωX − D (ω+ ), where C = π∗ (C ) and D = π∗ (D ). By applying π∗ to equation (33), one finds that J∗ (C) = δD. Since (ωX , ω + ) satisfies the integrality condition, it thus follows that C (ωX − J ∗ (θ + B)) ∈ Z.

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As an immediate consequence, we obtain the following main result of the section. Theorem 5.7. Let ( ⇒ M, ω + ) be an exact proper pre-quasi-symplectic J

groupoid, and (X → M, ωX ) a pre-Hamiltonian -space. Then there exists a compatible prequantization R → ⇒ M and L → X if and only if the pair (ωX , ω + ) satisfies the integrality condition of equation (27). Proof. Assume that (R → ⇒ M, θ +B) and (L → X, θL ) are a pair of compatible 2 ((R × X) , Z). prequantizations. By Corollary 4.7, we have ωX − J ∗ (θ + B) ∈ ZdR M • Hence (ωX , ω + ) satisfies the integrality condition according to Proposition 5.6. Conversely, assume that (ωX , ω + ) satisfies the integrality condition. Then ω + must be an integral cocycle. Let (R → ⇒ M, θ + B) be a prequantization, which always exists since is proper. Again according to Proposition 5.6, there exists 2 ( ) such that ω −J ∗ (θ +B)−J ∗ π ∗ + ∈ Z 2 ((R × X) , Z). a 2-cocycle + ∈ ZdR • X M • dR Since is proper, + is cohomologous to α + B0 , where α ∈ 1 () is a closed 1-form and B0 ∈ 2 (M). Then θ + B := (θ + π ∗ α) + (B + B0 ) is clearly also a pseudo2 ((R × X) , Z). From Corollary 4.7, it connection and ωX − J ∗ (θ + B ) ∈ ZdR M • J

follows that (X → M, ωX ) admits a compatible prequantization (L → X, θL ).

5.2 Integral quasi-Hamiltonian G-spaces In this subsection, G is a connected and simply-connected compact Lie group and 1 denotes the unit of G. We intend to study the case where is the AMM quasisymplectic groupoid. Assume that X is a G-space. There is a natural map i : H2 (X, Z) → H2 ((G × X)• , Z) induced by the inclusion C2 (X, Z) ⊂ C2 ((G×X)• , Z). The following lemma indicates that i is in fact an isomorphism. Lemma 5.8. If G is a connected and simply-connected Lie group, then the map i : H2 (X, Z) → H2 ((G × X)• , Z) is an isomorphism. Proof. This is a standard result. For completeness, we sketch a proof below. Let G → EG → BG be the usual G-bundle over the classifying space BG and XG = G\(EG × X). We have the fibration G → EG × X → XG . 2 The second term of the homology Leray–Serre spectral sequence is Ep,q = Hp (XG , Hq (G, Z)), i.e., the homology of XG with local coefficients in Hq (G, Z) (see [12]). Since G is simply-connected, we have H1 (G, Z) = H2 (G, Z) = 0 and 2 has the following form for 0 ≤ p ≤ 3 and 0 ≤ q ≤ 2: Ep,q .. .. .. .. . . . . 0 0 0 0 ··· 0 0 0 0 ··· H0 (XG , Z) H1 (XG , Z) H2 (XG , Z) H3 (XG , Z) · · ·

(34)


445

According to the Leray–Serre theorem, this spectral sequence converges to H∗ (EG × X, Z). It is clear from equation (34) that, in particular, we have H2 (EG × X, Z) ! H2 (XG , Z). Since EG is contractible, we get H2 (XG , Z) ! H2 (X, Z). The lemma now follows from the well-known isomorphism H2 ((G × X)• , Z) ! H2 (XG , Z).

Since H2 (g∗ , Z) = 0, Lemma 5.8 implies that H2 ((T ∗ G)• , Z) = 0.

(35)

Since any simply-connected Lie group G satisfies H2 (G, Z) = 0, we also have H2 ((G × G)• , Z) = 0.

(36)

Recall that the AMM quasi-symplectic groupoid is (G × G ⇒ G, ω + ) [6, 22], where G is a compact Lie group equipped with an ad-invariant nondegenerate symmetric bilinear form (·, ·). Here G × G ⇒ G is the transformation groupoid, where G acts on itself by conjugation, and ω and are defined as follows. Following [3], we denote by θ and θ¯ the left and right Maurer–Cartan forms on G, respectively, i.e., θ = g −1 dg and θ¯ = (dg)g −1 . Let ∈ 3 (G) denote the bi-invariant 3-form on G corresponding to the Lie algebra 3-cocycle 1 3 ∗ 12 (·, [·, ·]) ∈ ∧ g , i.e.,

=

1 1 ¯ (θ, [θ, θ]) = (θ¯ , [θ¯ , θ]), 12 12

(37)

and ω ∈ 2 (G × G) the 2-form 1 ω|(g,x) = − [(Adx pr ∗1 θ, pr ∗1 θ ) + (pr ∗1 θ, pr ∗2 (θ + θ¯ ))], 2

(38)

where (g, x) denotes the coordinate in G × G, and pr 1 and pr 2 : G × G → G are natural projections. It is known that ω + is an integral 3-cocycle. A triple (X, ωX , J ), where X is a manifold, ωX is a G-invariant 2-form on X and J : X → G is a smooth map, is a quasi-Hamiltonian G-space in the sense of [3] if (B1) the differential of ωX is given by dωX = J ∗ ; (B2) the map J satisfies ξˆ and

ωX =

1 ∗ J (ξ, θ + θ¯ ); 2

446


(B3) at each x ∈ X, the kernel of ωX is given by ker ωX = {ξˆ (x)|ξ ∈ ker(Ad J (x) +1)}, where ξˆ is the vector field on X associated to the infinitesimal action of ξ ∈ g on X. J

It is known [22] that these conditions are equivalent to (X → G, ωX ) being a Hamiltonian -space, where is the AMM quasi-symplectic groupoid (G × G ⇒ G, ω + ). In this case, the integrality can be described in simpler terms as indicated in the following. Proposition 5.9. Let be the AMM quasi-symplectic groupoid (G × G ⇒ G, ω +

), where G is a connected and simply-connected Lie group equipped with an J

ad-invariant nondegenerate symmetric bilinear form. Let (X → G, ωX ) be a quasi-Hamiltonian G-space. Assume that ω + is an integral 3-cocycle in 3 ((G × G) , Z). Then the pair (ω , ω + ) satisfies the integrality condition ZdR • X if and only if ∀C ∈ Z2 (X, Z) and D ∈ C3 (G, Z) such that dD = J∗ (C), ωX − ∈ Z. (39) C

D

Note that such D always exists for any C ∈ Z2 (X, Z). Proof. Note that we have the following commutating diagram of groupoid homomorphisms: i

X• → (G × X)• ↓J ↓J

(40)

J

G• → (G × G)• , where X• and G• are spaces X and G are considered as groupoids, while (G × X)• and (G × G)• are the transformation groupoids. Thus one direction is obvious. Conversely, according to equation (36), we have H2 ((G×G)• , Z) = 0. Therefore, Ker(J∗ ) = H2 ((G × X)• , Z). By Lemma 5.8, for any class C ∈ H2 ((G × X)• , Z), there exists C ∈ Z2 (X, Z) such that C = i∗ [C]. Since H2 (G, Z) = 0, there always exists D ∈ C3 (G, Z) such that J∗ (C) = dD. Hence J∗ (i∗ C) = i∗ (J∗ C) = i∗ dD = δ(i∗ D). Now it is clear that ∗ ∗ ωX − (ω + ) = i ωX − i (ω + ) = ωX − . i∗ C

i∗ D

C

D

The conclusion thus follows from Lemma 5.4.

C

D


447

Remark 5.10. Note that equation (39) coincides with the quantization condition of Alekseev–Meinrenken [2]. See also [16]. For the case of conjugacy classes, see [14, 15]. As an immediate consequence of Proposition 5.9, we have the following. Corollary 5.11. Let be the AMM quasi-symplectic groupoid (G × G ⇒ G, ω + ). Then 1 ∈ G, considered as a quasi-Hamiltonian G-space, satisfies the integrality condition. Let us consider the case of Example 4.3 where is the symplectic groupoid T ∗ G ⇒ g∗ . In this case, we recover a well-known result of Guillemin–Sternberg [10]. Proposition 5.12. Let be the symplectic groupoid (T ∗ G ⇒ g∗ , ω), where G is a connected and simply-connected Lie group. Let J : X → g∗ be a momentum map for a Hamiltonian G-space (X, ωX ) as in Example 4.3. The pair (ωX , ω) satisfies the integrality condition if and only if ωX is an integral 2-form. Proof. According to equation (35), we have H2 ((T ∗ G)• , Z) = 0. Therefore, for any C ∈ Z2 ((G × X)• , Z) there exists D ∈ C3 ((T ∗ G)• , Z) such that J∗ (C) = δD. By Lemma 5.8, we may assume that C ∈ Z2 (X, Z). Since H2 (g∗ , Z) = 0, we can assume that D ∈ C3 (g∗ , Z). Since = 0, the integrality condition of equation (27) thus reads C ωX ∈ Z.

In particular, a coadjoint orbit O ⊂ g∗ , endowed with the Kirillov–Kostant– Souriau symplectic structure ωO , satisfies the integrality condition if and only if ωO is an integral 2-form. 5.3 Integrality condition and Morita equivalence In general, a pre-quasi-symplectic groupoid may not be exact, as in the case of the AMM-quasi-symplectic groupoid for instance. In such a case, one must pass to a Morita-equivalent pre-quasi-symplectic groupoid in order to construct a prequantization. According to Theorem 4.12, Morita-equivalent quasi-(pre)symplectic groupoids yield equivalent momentum map theories in the sense that there is a bijection between their (pre)-Hamiltonian -spaces and the classical intertwiner spaces are independent of Morita equivalence [22]. More precisely, given a pre-quasi-symplectic groupoid ( ⇒ M, ω + ), where p

may not be exact, one can choose a surjective submersion N → M and consider the pullback groupoid [N] ⇒ N of ⇒ M via p. Then ([N] ⇒ N, p∗ ω + p∗ ) J

is again a pre-quasi-symplectic groupoid. Moreover, if (X → M, ωX ) is a preJN

Hamiltonian -space, then (XN → N, p∗ ωX ) is a pre-Hamiltonian [N]-space, where XN = X ×M N , and p : XN → X and JN : XN → N are the projections to the first and second components, respectively. The following proposition indicates that integrality condition is preserved under this pullback procedure.

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Lemma 5.13. The pair (ωX , ω + ) satisfies the integrality condition if and only if (p∗ ωX , p∗ ω + p ∗ ) satisfies the integrality condition. Proof. By abuse of notation, we use the same letter p to denote the groupoid homomorphisms from [N ] ×N XN ⇒ XN to ×M X ⇒ X, and from [N] ⇒ N to ⇒ M, both of which are Morita morphisms. For any C ∈ Z2 (([N]×N XN )• , Z) and D ∈ C3 ([N]• , Z) with J∗ (C ) = δD , we have p ∗ ωX − p ∗ (ω + ) = ωX − (ω + ), (41) C

(C )

D

C

D

(D )

and D = p∗ clearly satisfy J∗ (C) = δD. where C = p∗ Assume that the pair (ωX , ω + ) satisfies the integrality condition. Then equation (41) implies immediately that so too does the pair (p ∗ ωX , p∗ ω + p ∗ ). Conversely, if (p∗ ωX , p∗ ω + p ∗ ) satisfies the integrality condition, then ω + must be an integral cocycle. Now we have the commutative diagram: p∗

H2 (([N] ×N XN )• , Z) → H2 (( ×M X)• , Z) ↓ JN ∗ ↓ J∗ p∗ H2 ([N]• , Z) → H2 (• , Z), where the horizontal arrows are isomorphisms. Therefore, p∗ : H2 (([N] ×N XN )• , Z) → H2 (( ×M X)• , Z) induces an isomorphism from Ker(JN ∗ ) to Ker(J∗ ). This implies that any class in Ker(J∗ ) has a representative of the form C = p∗ (C ), where C = δD for some D ∈ C3 (([N] ×N XN )• , Z). Let D = p∗ (D ). By equation (41), we see that if the pair (p∗ ωX , p∗ ω + p ∗ ) satisfies the integrality condition then C ωX − D (ω + ) ∈ Z. By Lemma 5.4, we conclude that (ωX , ω + ) satisfies the integrality condition. Corollary 5.14. Let (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) be Moritaequivalent pre-quasi-symplectic groupoids. Assume that (F → G0 , ωF ) and (E → H0 , ωE ) are a pair of corresponding pre-Hamiltonian spaces. Then (ωF , ωG + G ) satisfies the integrality condition if and only if (ωE , ωH + H ) satisfies the integrality condition. Proof. It suffices to prove this assertion for a Morita morphism of pre-quasisymplectic groupoids. By Lemma 5.13, it remains to prove that the integrality condition is preserved by gauge transformations of the first type, which can be easily checked.

As a consequence, given a pre-quasi-symplectic groupoid ( ⇒ M, ω+ ), where p

may not be exact, one can choose a surjective submersion N → M such that p∗ ∈

3 (N) is exact and replace ( ⇒ M, ω + ) by a Morita-equivalent exact H pre-quasisymplectic groupoid ([N] ⇒ N, p∗ ω+p ∗ ). Usually, one takes N := Ui → M,


449

where U = (Ui ) is an H open cover of M. Then the pullback pre-quasi-symplectic groupoid is ([U] ⇒ Ui , ω|[U ] + |Ui ), where [U], as a manifold, can be H U identified with the disjoint union Uij . Lemma 4.7 guarantees that the integrality condition always holds no matter which surjective submersion (or open covering) N → M is taken as long as the initial pair (ωX , ω + ) satisfies the integrality condition, and therefore one can always construct a compatible prequantization. Applying the above discussion to the AMM quasi-symplectic groupoid (G×G ⇒ G, ω + ) and using Theorem 5.7, we are led to the following. J

Corollary 5.15. Let (X → G, ωX ) be a quasi-Hamiltonian G-space. The following are equivalent: H H (1) There exists H H a compatible prequantizationH Rij → (G × G)[U] ⇒ Ui and Li → X|Ui , where (G × G)[U] ⇒ Ui is the pullback quasi-symplectic groupoid of the AMM groupoid using any open covering of G such that ∀i, |Ui is an exact form. (2) The integrality condition of equation (39) holds. 5.4 Strong integrality condition Definition 5.16. Let ( ⇒ M, ω + ) be a pre-quasi-symplectic groupoid. A preHamiltonian -space (X → M, ωX ) is said to satisfy the strong integrality condition if (1) it satisfies the integrality condition; and 2 ( ) → H 2 (( × X) ) vanishes. (2) the map J ∗ : HdR • M • dR The following result follows from Theorem 5.7. Proposition 5.17. Let ( ⇒ M, ω + ) be an exact proper pre-quasi-symplectic J

J

groupoid, and (X → M, ωX ) a pre-Hamiltonian -space. Then (X → M, ωX ) satisfies the strong integrality condition if and only if for any prequantization of ( ⇒ M, ω + ), X admits a compatible prequantization. J

Proof. If (X → M, ωX ) satisfies the strong integrality condition, it is clear from Theorem 5.7 that X admits a compatible prequantization for any prequantization of ( ⇒ M, ω + ). Conversely, given any prequantization (R → ⇒ M, θ + B), J ∗ (θ + B) − ωX 2 ((R × X) , Z). Note that if θ + B is a pseudomust be an integral 2-cocycle in ZdR M • 2 ( ). Since the subset of integral classes connection, so is θ + B + π ∗ + ∀+ ∈ ZdR • 2 ((R × X) , Z) is discrete, then J ∗ (θ + B) − ω + J ∗ π ∗ + being an integral ZdR M • X cocycle for all + implies that [J ∗ ◦ π ∗ (+)] = 0. In other words, the map J ∗ ◦ π ∗ : 2 ( ) → H 2 ((R × X) ) is the zero map. Since R × X → × X ⇒ X HdR • M • M M dR 2 (( × X) ) → defines a trivial gerbe according to Proposition 2.3, the map π ∗ : HdR M • 2 ((R × X) ) is injective. From the identity J ∗ ◦ π ∗ = π ∗ ◦ J ∗ and the fact that HdR M • 2 ( ) → H 2 (( × X) ) must vanish.

π ∗ is injective, it follows that J ∗ : HdR • M • dR

450


The following proposition is an analogue of Corollary 5.14. Proposition 5.18. Let (G ⇒ G0 , ωG + G ) and (H ⇒ H0 , ωH + H ) be Moritaequivalent pre-quasi-symplectic groupoids. Assume that (F → G0 , ωF ) and (E → H0 , ωE ) are a pair of corresponding pre-Hamiltonian spaces. Then (ωF , ωG + G ) satisfies the strong integrality condition if and only if (ωE , ωH + H ) satisfies the strong integrality condition. Proof. By Corollary 5.14, we just have to check that Condition (2) in the definition of strong integrality condition is invariant under Morita equivalence. This follows immediately from the commutativity of the diagram 2 (G ) 2 (H ) ! HdR HdR • • ↓ ↓ 2 ((G × 2 HdR G0 F )• ) ! HdR ((H ×H0 E)• ),

where the horizontal arrows are the natural isomorphism between the de Rham cohomologies of two Morita-equivalent groupoids.

Remark 5.19. 2 ( , Z) = 0, then condition (2) in the definition of 1. If the groupoid satisfies HdR • the strong integrality is satisfied for any pre-Hamiltonian -space. In this case, a pre-Hamiltonian space satisfies the integrality condition if and only if it satisfies the strong integrality condition. 2. If G is a connected and simply-connected Lie group, then H2 ((G × G)• , Z) = 0. Therefore, any quasi-Hamiltonian G-space satisfying the integrality condition must satisfy the strong integrality condition.

The following proposition summarizes the results of this section. Proposition 5.20. Let ( ⇒ M, ω + ) be an exact, proper, pre-quasi-symplectic Jk

groupoid, and let (Xk → M, ωk ), k = 1, 2, be pre-Hamiltonian -spaces. Assume J1

J2

that (X1 → M, ω1 ) satisfies the integrality condition while (X2 → M, ω2 ) satisfies the strong integrality condition. Then there exists a prequantization of ( ⇒ M, ω +

) and compatible prequantizations of both X1 and X2 . Therefore, the classical intertwiner space X2 × X1 is quantizable. Applying this result to the case of the AMM quasi-symplectic groupoid, we have the following. Corollary 5.21. Let G be a connected and simply-connected compact Lie group J

equipped with an ad-invariant nondegenerate symmetric bilinear form, and (X → G, ωX ) a quasi-Hamiltonian G-space. Assume that ωX satisfies the integrality condition as in equation (39). Then the reduced symplectic manifold J −1 (1)/G is prequantizable, and the prequantization can be constructed H using the prequantization of the AMM quasi-symplectic groupoid (G × G)[U] ⇒ Ui (more precisely the pullback groupoid of the AMM quasi-symplectic groupoid ) together with a comH H patible prequantization of the Hamiltonian space ( X|Ui → Ui , ωX |Ui ), where U = (Ui )i∈I is some open covering of G such that |Ui is exact ∀i ∈ I .


451

6 Appendix We denote by CS 1 the canonical cycle in C1 (S 1 , Z) that generates H1 (S 1 , Z) = Z. If we consider CS 1 as an element of C2 (S•1 , Z), [CS 1 ] generates H2 (S•1 , Z) ! Z. For any point p in a manifold N , we denote by Cp the constant map from S 1 to {p} and consider it as an element of C1 (N, Z). Assume that R → ⇒ M is an S 1 -central extension of groupoids. For any m ∈ M, let Zm = fm∗ (CS 1 ) ∈ C2 (R• , Z),

(42)

where fm : S 1 → R is defined by equation (13). More generally, for any r ∈ R, let fr : S 1 → R be the map λ → λ · r, and set Zr = fr∗ (CS 1 ) − Cr ∈ C2 (R• , Z). Proposition 6.1. Let R → ⇒ M be an S 1 -central extension. Assume that M/ is connected. (1) The class [Zm ] ∈ H2 (R• , Z) does not depend on the choice of m ∈ M. Because of this, we will drop the subscript m and denote this class simply by [Z]. (2) For any r ∈ R, Zr is a cycle and [Zr ] = [Z]. (3) The natural map π∗ : H2 (R• , Z) → H2 (• , Z) is surjective. (4) Its kernel Ker(π∗ ) is generated by [Z]. (5) The following identity holds: θ = 1. Zm

Before we prove this proposition, we first need a lemma. Given any point p ∈ N , we will denote by Cp(k) the chain in Ck (N, Z) defined by the constant path k → {p}. π

Lemma 6.2. Let R → ⇒ M be an S 1 -central extension. (1) Any element E in C0 (R, Z) with π∗ (E) = 0 can be written of the form E = δD , where D ∈ C1 (R, Z) satisfies π∗ (D ) = 0. (2) π∗ : C• (R• , Z) → C• (• , Z) is a surjective map. (3) Any element in the kernel of π∗ : Hk (R• , Z) → Hk (• , Z) has a representative C ∈ Zk (R• , Z) with π∗ (C) = 0. (4) Any element C in C0 (R2 , Z) with π∗ (C) = 0 is of the form C = dD , where D ∈ C1 (R2 , Z) satisfies π∗ (D ) = 0. (5) For any cycle C ∈ C1 (R, Z) such that δC = 0 and π∗ (C ) = 0, we have [C ] = ki [Zri ] i∈I

for some finite set I , ki ∈ Z and ri ∈ R.

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Proof. (1) The kernel of π∗ : C0 (R, Z) → C0 (, Z) is generated by elements of the π form p − q, where p and q are two points in the same fibre of R → . Hence, it suffices to prove the claim for such a generator. Let D : 1 → R be a path in the fiber π −1 (p) satisfying dD = p − q. Set D = D −Cp(1) . Clearly, the identities dD = p −q and π∗ (D ) = 0 hold. Moreover, from π∗ (D ) = 0, it follows that ∂D = s∗ π∗ (D ) − t∗ π∗ (D ). Hence δD = p − q (2) Since the projections π : Rk → k are surjective submersions with fibers isomorphic to k-dimensional torus, all the maps π∗ : Cl (Rk , Z) → Cl (k , Z) are onto for all k, l ∈ N. (3) Let C ∈ Zk (R• , Z) be a cycle with π∗ [C ] = 0. By definition, there exists D ∈ Ck+1 (• , Z) such that δD = π∗ (C ). By (2), there exists D in Ck+1 (R• , Z) such that π∗ (D ) = D. Set C := C − δD . We have [C] = [C ] and π∗ (C) = 0. (4) The kernel of π∗ : C0 (R2 , Z) → C0 (2 , Z) is generated by elements of the form p − q, where p and q are two points on the same fiber of R2 → 2 . It thus suffices to show this property for such generators. Let D : 1 → R2 be a path in the fiber over π(p) such that dD = p − q. Let D = D − Cp(1) . Thus π∗ (D ) = π∗ (D − Cp(1) ) = Cπ(p)(1) − Cπ(p)(1) = 0

and

dD = p − q.

(5) For simplicity, we call those chains in C1 (R, Z) of the form C − Cp(1) fibered 1-chains, where p ∈ R is a point and C : 1 → π −1 (π(p)) is a path in the fiber through the point p. Any fibered 1-chain is in the kernel of π∗ and hence lies in the kernel of ∂. If a fibered 1-chain E in a given fiber satisfies dE = 0, then [E] = k[Zr ] for some r ∈ R and k ∈ Z. As a consequence, if a linear combination of fibered 1-chains F is a cycle in C1 (R, Z), then it is clear that [F ] = i∈I ki [Zri ] for some finite set I , ki ∈ Z and ri ∈ R. Now the kernel of π∗ : C1 (R, Z) → C1 (, Z) is generated by elements of the form C0 − C1 , where Ci , i = 0, 1, are paths 1 → R satisfying π∗ (C0 ) = π∗ (C1 ). Thus there is a map γ : 1 → S 1 such that C0 (t) = γ (t) · C1 (t) ∀t ∈ 1 . Let γ˜ : [0, 1] × 1 → S 1 be a map with γ˜ (0, t) = 1 and γ˜ (1, t) = γ (t). Let us define two maps D1 and Dˆ : [0, 1] × 1 → R by D1 (s, t) = γ˜ (s, t) · C0 (t) and ˆ We have π∗ (D) = 0 and therefore ∂D = 0. ˆ t) = C0 (t). Set D := D1 − D. D(s, Moreover, by construction, C0 −C1 +δD = C0 −C1 +dD is the sum of two 1-fibered chains: one in the fiber through C0 (0) and another in the fiber through C0 (1). The conclusion thus follows.

Proof of Proposition 6.1. (1), (2) It is clear that if m and n are in the same connected component of M, then [Zm ] = [Zn ]. Now by the definition of Zr , we have dZr = d(fr∗ (CS 1 )) − dCr = 0, s∗ (Zr ) = s∗ (fr∗ (CS 1 ) − Cr ) = Cs(r) − Cs(r) = 0, and


453

t∗ (Zr ) = t∗ (fr∗ (CS 1 ) − Cr ) = Ct (r) − Ct (r) = 0. Therefore, δ(Zr ) = 0. Consider the map D : S 1 → R2 defined by λ → (fr (λ), ft (r) (λ−1 )). We have dD = 0 and ∂D = fr∗ (CS 1 ) − Cr − ft (r)∗ (CS 1 ). Hence we have [Zr ] = [Zt (r) ] ∀r ∈ R. Similarly, we have [Zr ] = [Zs(r) ] ∀r ∈ R. Since M/ is connected, (1) and (2) follow. (3) Let C ∈ Z2 (• , Z) be any 2-cycle. According to Lemma 6.2 (2), there exists D ∈ C2 (R• , Z) with π∗ (D) = C. In general, δD = 0. However since the restriction of π to M is the identity map, we have ∂D1 − dD2 = 0 and thus δD = ∂D0 − dD1 , where D = D0 + D1 + D2 , Di ∈ Ci (R2−i , Z). Therefore, δD is an element of C0 (R, Z) and π∗ (δD) = δπ∗ (D) = δC = 0. By Lemma 6.2(1), there exists D ∈ C2 (R• , Z) with π∗ (D ) = 0 and δD = δD. Therefore, it follows that D − D is a cycle in Z2 (R• , Z) and π∗ ([D − D ]) = [π∗ (D)] − [π∗ (D )] = [C] − [0] = [C]. (4) According to Lemma 6.2 (3), any class in Ker(π∗ ) has a representative C such that π∗ (C) = 0 and therefore is of the form C0 + C1 , where C0 ∈ C0 (R2 , Z) and C1 ∈ C1 (R, Z) satisfy π∗ (C0 ) = 0 and π∗ (C1 ) = 0. According to Lemma 6.2 (4), there exists D ∈ C1 (R2 , Z) with π∗ (D ) = 0 such that C0 = dD . Consider now C = C − δD ∈ C1 (R, Z). We have δC = δC − δ 2 D = 0,

[C ] = [C],

According to Lemma 6.2(5), we have ki [Zri ] [C ] =

π∗ (C ) = 0.

(43)

i∈I

for some finite set I , ki ∈ Z and ri ∈ R. From equation (43), it follows that [C] = [C ] = i∈I ki [Zri ]. By Lemma 6.1 (2), we have [C] = ( i∈I ki )[Z]. (5) This holds because θ is a connection 1-form of the S 1 -principal bundle R → .

Acknowledgments The second author would like to thank the Erwin Schrödinger Institute and the University of Geneva for their hospitality while work on this project was being done. We would like to thank Anton Alekseev, Kai Behrend, Eckhard Meinrenken, and Jim Stasheff for useful discussions.

References [1] Alekseev, A., On Poisson actions of compact Lie groups on symplectic manifolds, J. Differential Geom., 45 (1997), 241–256. [2] Alekseev, A., and Meinrenken, E., private communication. [3] Alekseev, A., Malkin, A., and Meinrenken, E., Lie group valued moment maps, J. Differential Geom., 48 (1998), 445–495.

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[4] Behrend, K., and Xu, P., S 1 -bundles and gerbes over differentiable stacks, C. R. Acad. Sci. Paris Sér. I, 336 (2003), 163–168. [5] Behrend, K., and Xu, P., Differential stacks and gerbes, in preparation. [6] Behrend, K., Xu, P., and Zhang, B., Equivariant gerbes over compact simple Lie groups, C. R. Acad. Sci. Paris Sér. I, 336 (2003), 251–256. [7] Bursztyn, H., Crainic, M., Weinstein, A., and Zhu, C., Integration of twisted Dirac brackets, Duke Math. J., 123-3 (2004), 549–607. [8] Dupont, L., Curvature and Characteristic Classes, Lecture Notes in Mathematics, Vol. 640, Springer-Verlag, New York, 1978. [9] Ginzburg, V., and Weinstein, A., Lie–Poisson structure on some Poisson Lie groups, J. Amer. Math. Soc., 5 (1992), 445–453. [10] Guillemin, V., and Sternberg, S., Geometric quantization and multiplicities of group representations, Invent. Math., 67 (1982), 515–538. [11] Laurent-Gengoux, C., Tu, J.-L., and Xu, P., Chern–Weil map and characteristic classes of principal G-bundles over groupoids, math.DG/0401420. [12] Mc Cleary, J., A User’s Guide to Spectral Sequences, 2nd ed., Cambridge Studies in Advanced Mathematics, Vol. 2, Cambridge University Press, Cambridge, UK, 2000. [13] Meinrenken, E., Symplectic surgery and the SpinC -Dirac operator, Adv. Math., 134 (1998), 240–277. [14] Meinrenken, E., The basic gerbe over a compact simple Lie group, Enseign. Math. (2), 49 (2003), 307–333. [15] Mohrdieck, S., and Wendt, R., Integral conjugacy classes of compact Lie groups, Manuscripta Math., 113 (2004), 531–547. [16] Shabhazi, Z., Ph.D. thesis, Department of Mathematics, University of Toronto, Toronto, 2004. [17] Spanier, E., Algebraic Topology, Springer-Verlag, New York, 1981. [18] Tu, J.-L., Xu, P., and Laurent-Gengoux, C., Twisted K-theory of differentiable stacks, Ann. Sci. École Norm. Sup., to appear; math.KT/0306138. [19] Weinstein, A., and Xu, P., Extensions of symplectic groupoids and quantization, J. Reine Angew. Math., 417 (1991), 159–189. [20] Xu, P., Morita equivalent symplectic groupoids, in Dazord, P., and Weinstein, A., eds., Symplectic Geometry, Groupoids, and Integrable Systems (Berkeley, CA, 1989), Mathematical Sciences Research Institute Publications, Vol. 20, Springer-Verlag, New York, 1991, 291–311. [21] Xu, P., Classical intertwiner spaces and quantization, Comm. Math. Phys., 164 (1994), 473–488. [22] Xu, P., Momentum map and Morita equivalence, J. Differential Geom., to appear; math.SG/0307319.

Duality and triple structures Kirill C. H. Mackenzie Department of Pure Mathematics University of Sheffield Sheffield S3 7RH UK [email protected] Dedicated to Alan Weinstein on the occasion of his sixtieth birthday. Abstract. We recall the basic theory of double vector bundles and the canonical pairing of their duals, introduced by the author and by Konieczna and Urbański. We then show that the relationship between a double vector bundle and its two duals can be understood simply in terms of an associated cotangent triple vector bundle structure. In particular, we show that the dihedral group of the triangle acts on this triple via forms of the isomorphisms R , introduced by the author and Ping Xu. We then consider the three duals of a general triple vector bundle and show that the corresponding group is neither the dihedral group of the square nor the symmetry group on four symbols.

Double structures first appeared in Poisson geometry with Alan’s groundbreaking work on symplectic groupoids [Coste, Dazord, and Weinstein 1987], [Weinstein 1987] and Poisson groupoids [Weinstein 1988]. The most fundamental example of a symplectic groupoid, the cotangent groupoid T ∗ G of an arbitrary Lie groupoid G , introduced in [Coste et al. 1987], is a groupoid object in the category of vector bundles. An arbitrary Poisson Lie group can be integrated to a symplectic double groupoid [Lu and Weinstein 1989]. At a simpler level, a Poisson structure on a vector bundle is linear [Courant 1990] if and only if the associated anchor is a morphism of certain double vector bundles. All these phenomena involve doubles in the categorical sense: taking S to denote, for example, “vector bundle’’ or “Lie groupoid,’’ a double S is an S object in the category of all S . (Groupoid objects in the category of vector bundles, named VBgroupoids by Pradines [1988], may be regarded as double groupoids of a special type.) More generally, multiple S structures are the n -fold extension of this notion of double. The key link between Poisson geometry and double structures lies in properties of the Poisson anchor. If a Poisson manifold P is a vector bundle on base M , then the Poisson structure is linear if and only if π # : T ∗ P → T P is a morphism of double vector bundles. If P is instead a Lie groupoid on base M , then the groupoid

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is a Poisson groupoid if and only if π # is a morphism of VB-groupoids. Thus the Poisson anchor naturally appears as a map of double structures, and indeed many of the surprising basic features of Poisson and symplectic groupoids are not really so much consequences of Poisson or symplectic geometry as consequences of the duality properties of the associated double structures. This point of view is developed further in [Mackenzie 2004]; in particular, the theory of Poisson groupoids may be developed entirely in terms of groupoid theory and double structures of various kinds. The present paper is concerned with the duality of double and higher multiple vector bundles. A double vector bundle has two duals which are themselves in duality and we show here that the various combinations of the two dualization operations gives rise to the dihedral (or symmetric) group of order six. We show in Section 5 and Section 6 that a double vector bundle and its two duals form the three lower faces of a triple vector bundle, the opposite vertex of which is the cotangent of the double space. This encapsulates and makes symmetric the relations between a double vector bundle and its duals, which can otherwise seem rather involved. One may think of three double vector bundles with a common vertex and appropriate pairings as constituting a two (sic) dimensional version of the familiar notion of pairing of vector bundles; we call this a cornering. In Section 7 we consider the process of dualizing the structures in a triple vector bundle. This may appear to be a routine extension of the double case, but we show that the group of dualization operations here is not the dihedral group of the square, or the symmetric group on four symbols, but a group of order 72. This appears to demonstrate that the behaviour of duality for n -fold vector bundles may be a less routine extension of the double case than one might have expected. In the final Section 8, we formulate some general principles which we believe do hold for general multiple vector bundles. The study of general double vector bundles was begun by Pradines [1974], although the case of the tangent double of an ordinary vector bundle (1.3) had been used in connection theory since the late 1950s. More than a decade later, Pradines [1988] introduced the dualization process for VB-groupoids; in the case of double vector bundles this is the duality construction presented here in Section 3. Theorem 3.2 is from [Mackenzie 1999] and was also found by Konieczna and Urban´ ski [1999]. The idea of deriving the pairing (17) from the cotangent triple was noted in [Mackenzie 2002]. The results of Section 4 first appeared in the paper [Mackenzie and Xu 1994] of Ping Xu and myself. They are here obtained as a consequence of the general duality of double vector bundles. An expanded account of the double case may be found in [Mackenzie 2004].

1 Double vector bundles Definition 1.1. A double vector bundle (D; A, B; M) is a system of four vector bundle structures

Duality and triple structures

457

qBD D −−−−−−−−→ B ⏐ ⏐ qAD ?

⏐ ⏐ ? qB

(1)

A −−−−−−−−→ M qA in which D has two vector bundle structures, on bases A and B , which are themselves vector bundles on M , such that each of the structure maps of each vector bundle structure on D (the bundle projection, addition, scalar multiplication and the zero section) is a morphism of vector bundles with respect to the other structure. We refer to A and B as the side bundles of D , and to M as the double base. In the two side bundles the addition, scalar multiplication and subtraction are denoted by the usual symbols + , juxtaposition, and − . We distinguish the two zero sections, B B writing 0A : M → A , m → 0A m , and 0 : M → B , m → 0m . We may denote D an element d ∈ D by (d; a, b; m) to indicate that a = qA (d) , b = qBD (d) , m = qB (qBD (d)) = qA (qAD (d)). The notation qAD is clear; when the base of the bundle is the double base we write A. qA , for example, rather than qM In the vertical bundle structure on D with base A the vector bundle operations are denoted + , A. , − , with 0A : A → D , a → 0A a , for the zero section. Similarly, A A in the horizontal bundle structure on D with base B , we write + , B. , − and B B A B 0B : B → D , b → 0B b . For m ∈ M the double zero 00A = 00B is denoted m or m

m

02m . The two structures on D , namely (D, qBD , B) and (D, qAD , A) , will occasionally B and D A , respectively. be denoted D In dealing with general double vector bundles such as (1), we thus usually label objects and operations in the two structures on D by the symbol for the base over which they take place. The words “horizontal’’ and “vertical’’ may be used as an alternative, but need to be referred to the arrangement in the diagram (1) or the sequence in (D; A, B; M). When considering examples in which A = B , the words “horizontal’’ and “vertical’’ become necessary, and we use H and V as labels to distinguish the two structures on D . Although the concept of double vector bundle is symmetric, most examples are not; in the sequel it will be important to distinguish between (1) and its flip in Figure 1(a), in which the arrangement of the two structures is reversed. In such processes it is not the absolute arrangement which is significant, but the distinction between whichever arrangement is taken at the start and its flip. The condition that each addition in D is a morphism with respect to the other is (d1 + d2 ) + (d3 + d4 ) = (d1 + d3 ) + (d2 + d4 ) B

A

B

A

B

A

(2)

for quadruples d1 , . . . , d4 ∈ D such that qBD (d1 ) = qBD (d2 ) , qBD (d3 ) = qBD (d4 ) , qAD (d1 ) = qAD (d3 ) , and qAD (d2 ) = qAD (d4 ) . Next,

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K. C. H. Mackenzie

D

flip

D qA −→ A

⏐ D ⏐ qB ?

T (q) T E −→ T M ⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

B −→ M

E −→ M

(a)

(b) Fig. 1.

t A. (d1 + d2 ) = t A. d1 + t A. d2 , B B

(3)

for t ∈ R and d1 , d2 ∈ D with qBD (d1 ) = qBD (d2 ) ; similarly, t B. (d1 + d2 ) = t B. d1 + t B. d2 , A

A

(4)

for t ∈ R and d1 , d2 ∈ D with qAD (d1 ) = qAD (d2 ) . The two scalar multiplications are related by t A. (u B. d) = u B. (t A. d), (5) where t, u ∈ R and d ∈ D . Lastly, for compatible a, a ∈ A and compatible b, b ∈ B , and t ∈ R ,

and

A + A 0A a+a = 0a B 0a ,

. A 0A ta = t B 0a ,

(6)

B + 0B 0B b+b = 0b b ,

. B 0B tb = t A 0b .

(7)

A

Equations (2)–(7) are known as the interchange laws. Definition 1.2. A morphism of double vector bundles (ϕ; ϕA , ϕB ; f ) : (D; A, B; M) → (D ; A , B ; M ) consists of maps ϕ : D → D , ϕA : A → A , ϕB : B → B , f : M → M , such that each of (ϕ, ϕB ), (ϕ, ϕA ), (ϕA , f ), and (ϕB , f ) is a morphism of the relevant vector bundles. If M = M and f = id M , we say that ϕ is over M ; if, further, A = A and ϕA = id A , we say that ϕ is over A or preserves A . If A = A and B = B and both ϕA and ϕB are identities, we say that ϕ preserves the side bundles. Example 1.3. For an ordinary vector bundle (E, q, M) , applying the tangent functor to each of the bundle operations yields the tangent prolongation vector bundle (T E, T (q), T M). The zero section is T (0) : T M → T E . We denote the addition by + + and the scalar multiplication and subtraction by and . Together with the standard structure (T E, pE , E) , we have a double vector bundle (T E; E, T M; M), shown in Figure 1(b). There is no preferred arrangement for the side bundles of T E .

.


459

Example 1.4. Let A, B and C be any three vector bundles on the one base M , and write D for the pullback manifold A ×M B ×M C over M . Then D may be regarded as the direct sum qA! B ⊕ qA! C over A , and as the direct sum qB! A ⊕ qB! C over B , and with respect to these two structures, D is a double vector bundle with side bundles A and B . We call this the trivial double vector bundle over A and B with core C . It is tempting, but incorrect, to denote it by A ⊕ B ⊕ C . Example 1.5. A double vector bundle (D; A, B; M) may be pulled back over both of its side structures simultaneously. Suppose given vector bundles (A , qA , M ) and (B , qB , M ) and morphisms ϕ : A → A and ψ : B → B , both over a map f : M → M . Let D denote the set of all (a , d, b ) such that ϕ(a ) = qAD (d) , ψ(b ) = qBD (d) and qA (a ) = qB (b ) . Then, with the evident structures, (D ; A , B ; M ) is a double vector bundle and the projection D → D is a morphism over ϕ , ψ , and f . Further examples follow later in the paper.

2 The core and core sequences Until Example 2.2, consider a fixed double vector bundle (D; A, B; M). Each of the bundle projections is a morphism with respect to the other structure and so has a kernel (in the ordinary sense); denote by C the intersection of the two kernels: D A C = {c ∈ D | ∃m ∈ M such that qBD (c) = 0B m , qA (c) = 0m }.

This is an embedded submanifold of D . We will show that it has a well-defined vector bundle structure with base M , projection qC which is the restriction of qB ◦ qBD = qA ◦ qAD and addition and scalar multiplication which are the restrictions of either of the operations on D . Note first that the two additions coincide on C since c + c = (c + m ) + (m + c ) = (c + m ) + (m + c ) = c + c , B

c, c

A

B

A

B

A

B

A

(c ) ,

for ∈ C with qC (c) = qC using (2). From this it follows that t B. c = t A. c for integers t , and consequently for rational t , and hence for all real t by continuity. It will often be helpful to distinguish between c ∈ C , regarding C as a distinct vector bundle, and the image of c in D , which we will denote by c . Given c, c ∈ C with qC (c) = qC (c ) there is a unique c + c ∈ C with c = c + c , c + c = c + B A and given t ∈ R there is a unique tc ∈ C such that tc = t B. c = t A. c. It is now easy to prove that (C, qC , M) is a (smooth) vector bundle, which we call the core of (D; A, B; M).

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Theorem 2.1. There is an exact sequence (q D )! τA A −−B−2 qA! B qA! C >−−−> D

(8)

of vector bundles over A , and an exact sequence (q D )! τB B −−A−2 qB! A qB! C >−−−> D

(9)

+ of vector bundles over B , where the injections are τA : (a, c) → 0A a B c and D D B ! ! τB : (b, c) → 0b + c , respectively, and (qB ) and (qA ) denote the maps induced A D D by qB and qA into the pullback bundles. Proof. Take a ∈ Am , c ∈ Cm , where m ∈ M . Then both 0A a and c project under D D B A + qB to 0m . So 0a c is defined and also projects under qB to 0B m . That τA is linear B over A follows from the interchange laws. D Suppose that d ∈ D has qBD (d) = 0B m for some m ∈ M . Write a = qA (d) . D A A B A − − − Then d B 0a is defined and qB (d B 0a ) = 0m . On the other hand, q (d B 0A a)= A ∈ C . This establishes the exactness of (8). The proof of − 0 a − a = 0A . So d m m a B (9) is similar.

We refer to (8) as the core sequence of D over A , and to (9) as the core sequence of D over B . If (ϕ; ϕA , ϕB ; f ) : (D; A, B; M) → (D ; A , B ; M ) is a morphism of double vector bundles, then ϕ : D → D maps C into C , the core of D . It is clear that the restriction, ϕC : C → C , is a morphism of the vector bundle structures on the cores over f : M → M . Examples 2.2. For E an ordinary vector bundle, consider the tangent double vector bundle (T E; E, T M; M). The kernel of T (q) consists of the vertical tangent vectors and the kernel of pE consists of the vectors tangent along the zero section; their intersection is naturally identified with E itself. For clarity we distinguish X ∈ E from the core element X ∈ T E . The injection map for T E over E is the map τ which sends (X, Y ) ∈ Em × Em to the vector in Em which has tail at X and is parallel to Y . In terms of the prolongation structure, τ (X, Y ) = 0X + + Y . The injection map over T M is υ : (x, Y ) → T (0)(x) + Y . For ϕ : E → E a morphism of vector bundles over f : M → M , the morphism T (ϕ) of the tangent double vector bundles induces ϕ : E → E on the cores. In the case where ϕ and f are surjective submersions, the vertical subbundles form a double vector subbundle (in an obvious sense) (T ϕ E; E, T f M; M) of T E , the core of which is the kernel (in the ordinary sense) of ϕ . The trivial double vector bundle A ×M B ×M C of 1.4 has core C .


461

3 Duals of double vector bundles Throughout this section we consider a double vector bundle as in (1), with core bundle C . We will show that dualizing either structure on D leads again to a double vector bundle; in the case of the dual of the structure over A we denote this by D ×A qA×A

qC×∗A −−−−−−−−→ C ∗

⏐ ⏐ ?

⏐ ⏐ ? qC ∗

(10)

−−−−−−−−→ M. qA

A

Here C ∗ is the ordinary dual of C as a vector bundle over M . We denote the dual of D as a vector bundle over A by D × A . (We will later modify this notation for cases in which A and B are identical.) The vertical structure in (10) is the usual dual of the bundle structure on D with base A , and qC ∗ : C ∗ → M is the usual dual of qC : C → M. The additions and scalar multiplications in the side bundles of (10) will be denoted by the usual plain symbols as before. In the two structures on D × A we write + , A. , − and A A + , . , − . The zero of D × A above a ∈ A is denoted 0 ×A . C∗

C∗

C∗

a

The unfamiliar projection qC×∗A : (D × A) → C ∗ is defined by + c, qC×∗A (), c = , 0A a B

(11)

where c ∈ Cm , : (qAD )−1 (a) → R and a ∈ Am . The addition +∗ in D × A → C ∗ C is defined by +∗ , d + d = , d + , d (12) C

B

That this is well defined depends strongly on the condition qC×∗A () = qC×∗A (#). Similarly, define t .∗ , t . d = t, d, C

B

qA×A (). for t ∈ R and d ∈ D with qAD (d) = ∗ is denoted The zero above κ ∈ Cm 0κ×A and is defined by + c = κ, c, 0κ×A , 0B b A

(13)

∗ is where b ∈ Bm , c ∈ Cm . The core element ψ corresponding to ψ ∈ Bm

+ ψ, 0B b A c = ψ, c. It is straightforward to verify that (10) is a double vector bundle and that its core is B ∗ . We call (10) the vertical dual or dual over A of (1).

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As for any double vector bundle, there are exact sequences A ! (qC× ∗ ) σA qA! B ∗ >−−−> D × A −−−2 qA! C ∗ ,

(14)

of vector bundles over A and (qA×A )! σC ∗ qC! ∗ B ∗ >−−−> D × A −−−2 qC! ∗ A,

(15)

of vector bundles over C ∗ . Here the two injections are given by ×A

σA (a, ψ) = 0a

×A

σC ∗ (κ, ψ) = 0κ

+ ψ,

C∗

+ ψ, A

where a ∈ A, ψ ∈ B ∗ , κ ∈ C ∗ . It is easily seen that σA (a, ψ), d = ψ, qBD (d) for d ∈ D and so σA is precisely the dual of (qBD )! . It is clear from the definition of qC×∗A that (qC×∗A )! = τV∗ . Thus (14) is precisely the dual of the core exact sequence (8). For the sequence over C ∗ we have + c = κ, c + ψ, b σC ∗ (κ, ψ), 0B b A

∗ , ψ ∈ B∗ , x ∈ B , c ∈ C . for κ ∈ Cm m m m The proof of the following result is straightforward. In Figure 2 and in similar figures in future, we omit arrows which are the identity.

Proposition 3.1. Consider a morphism of double vector bundles, as in Figure 2(a), which preserves the horizontal side bundles, and which has core morphism ϕC : C → C , where C is the core of D . Dualizing ϕ as a morphism of vector bundles over A, we obtain a morphism ϕ × A of double vector bundles over A and ϕC∗ , as in Figure 2(b), with core morphism ϕB∗ . This completes the description of the vertical dual of (1). There is of course also a horizontal dual qB×B × D B −−−−−−−−→ B qC×∗B

⏐ ⏐ ? C∗

⏐ ⏐ ? qB

(16)

−−−−−−−−→ M, qC ∗

with core A∗ → M , defined in an analogous way. The following result is an entirely new phenomenon, arising from the double structures.


D × A −→ (C )∗

D −→ B

H H ⏐ HH ⏐ H ϕB ϕH ⏐ ⏐ HH ? ? H j H H j H

A −→ M

⏐ ⏐ ?

D −→ B ⏐ ⏐ ?

A

⏐ ⏐ ?

H

H ⏐

H

H ϕC∗ H HH HH j H j

H⏐ ϕ × A ?H −→ M

463

D × A −→ C ∗ ⏐ ⏐ ?

⏐ ⏐ ?

A −→ M

A

−→ M

(a)

(b) Fig. 2.

Theorem 3.2 ([Mackenzie 1999], [Konieczna and Urbanski 1999]). There is a ´ natural (up to sign) duality between the bundles D × A and D × B over C ∗ given by , # = , dA − #, dB ,

(17)

where ∈ D × A, # ∈ D × B have qC×∗A () = qC×∗B (#) and d is any element of D with qAD (d) = qA×A () and qBD (d) = qB×B (#). Each of the pairings on the RHS of (17) is a canonical pairing of an ordinary vector bundle with its dual, the subscripts there indicating the base over which the pairing takes place. Proof. Let and # have the forms (; a, κ; m) and (#; κ, b; m) . Then d must have the form (d; a, b; m) . If d also has the form (d ; a, b; m) , then there is a + c ∈ Cm such that d = d + ( 0A a B c) , and so A , dA = , d A + κ, c + c) and so ( 0B by (11). By the interchange law (2) we also have d = d + b B A

#, dB = #, d B + κ, c. Thus (17) is well defined. To check that it is bilinear is routine. It remains to prove that it is nondegenerate. Suppose , given as above, is such that , # = 0 for all # ∈ (qC×∗B )−1 (κ). Take any ϕ ∈ A∗m and consider # = 0κ×B + ϕ . Then, taking d = 0A a we find B , dA = 0 and #, dB = ϕ, a. Thus ϕ, a = 0 for all ϕ ∈ A∗m and so × a = 0A m . It therefore follows from the horizontal exact sequence for D A that = 0κ×A + ψ A

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K. C. H. Mackenzie

∗ . Now taking any c ∈ C and defining d = + for some ψ ∈ Bm 0B m b A c , we find that

, dA = κ, c + ψ, b

and

#, dB = κ, c.

So ψ, b = 0 for all b ∈ Bm , since a suitable # exists for any given b . It follows ∗ and so is indeed the zero element over κ . Thus the pairing (17) that ψ = 0 ∈ Bm is nondegenerate.

Note several special cases: 0κ×B = 0, 0κ×A ,

0b×B = 0, 0a×A ,

0a×A , ϕ = −ϕ, a, ψ, 0b×B = ψ, b, ψ, ϕ = 0, A B × × , 0κ + ϕ = −ϕ, a, 0κ + ψ, # = ψ, b, A

B

(18) (19) (20)

where b ∈ B , a ∈ A , ϕ ∈ A∗ , ψ ∈ B ∗ and we have (#; κ, b; m) ∈ D × B and (; a, κ; m) ∈ D × A . Although we have proved that D × A and D × B are dual as vector bundles over ∗ C , we have not yet considered the relationships between the other structures present. This is taken care of by the following result, the proof of which is straightforward. Proposition 3.3 ([Mackenzie 1999]). Let (D; A, B; M) and (E; A, W ; M) be double vector bundles with a side bundle A in common, and with cores C and L, respectively. Suppose given a nondegenerate pairing , of D over A with E over A, and two further nondegenerate pairings, both denoted , , of B with L and of C with W , such that (i) for all b ∈ B , ∈ L, 0B b , = b, ; 0W (ii) for all c ∈ C , w ∈ W , c, w = c, w ; (iii) for all c ∈ C , ∈ L, c, = 0; (iv) for all d1 , d2 ∈ D , e1 , e2 ∈ E such that qBD (d1 ) = qBD (d2 ), E (e ) = q E (e ), q D (d ) = q E (e ) , q D (d ) = q E (e ), we have qW 1 W 2 A 1 A 1 A 2 A 2 d1 + d2 , e1 + e2 = d1 , e1 + d2 , e2 ; B W (v) for all d ∈ D , e ∈ E such that qAD (d) = qAE (e) and all t ∈ R , we have t B. d, t W. e = t d, e . ( In all the above conditions we assume the various elements of the side bundles lie in compatible fibres over M.) Then the map Z : D → E × A defined by Z(d), eA = d, e is an isomorphism of double vector bundles, with respect to id : A → A and the isomorphisms B → L∗ and C → W ∗ induced by the pairings in (i) and (ii). A pairing , satisfying the conditions of Proposition 3.3 is called a pairing of the double vector bundles. Applying this result to the pairing (17) of D × A and D × B , we find that the induced pairing of B with B ∗ is the standard one, but that of A∗ with A is the negative of the standard pairing. Hence the signs in the following result are unavoidable.


465

Corollary 3.4. The pairing (17) induces isomorphisms of double vector bundles ZA : D × A → D × B × C ∗ ,

ZA (), #C ∗ = , # ,

ZB : D × B → D × A× C ∗ ,

ZB (#), C ∗ = , #

with (ZA ) × C ∗ = ZB . Both isomorphisms induce the identity on the sides C ∗ → C ∗ . ZA is the identity on the cores B ∗ → B ∗ , and induces − id on the side bundles A → A. ZB is the identity on the side bundles B → B , and induces − id on the cores A∗ → A∗ . Example 3.5. Consider a trivial double vector bundle D = A ×M B ×M C. Let = (a, ψ, κ) be an element of D × A = A×M B ∗ ×M C ∗ and let # = (ϕ, b, κ) be an element of D × B . Then taking any d = (a, b, c) ∈ D , we find that , # = ψ, b − ϕ, a. The associated maps are given by ZA : A ×M B ∗ ×M C ∗ → A ×M B ∗ ×M C ∗ , ZB : A∗ ×M B ×M C ∗ → A∗ ×M B ×M C ∗ ,

(a, ψ, κ) → (−a, ψ, κ); (ϕ, b, κ) → (−ϕ, b, κ).

The following result is essentially equivalent to Theorem 3.2, but deserves independent statement. Theorem 3.6. For any double vector bundle (D; A, B; M) there is a canonical isomorphism Q from D to the flip of (D × A × C ∗ × B) which preserves the side bundles A and B and is − id on the cores C . Proof. Let $ = ZA × A be the dualization of ZA over A . Denote by F : D → D d , and define Q = (F ◦ $)−1 .

the map d → − B There are now three operations on double vector bundles: taking the vertical dual, denoted by V , taking the horizontal dual, denoted H , and the operation V H V which by Theorem 3.6 combines the flip and reversal of the sign on the core; we denote this by P . We have V 2 = H 2 = P 2 = I , the identity operation and, by the same method as Theorem 3.6, H V H = P . The group generated by V , H and P therefore has elements I,

V,

HV,

V HV = P,

and is the dihedral group

3

H V H V = H P = V H,

V H V H V = H, (21) of the triangle, or the symmetric group S3 .

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K. C. H. Mackenzie

4 Duals of T E Consider the tangent prolongation double vector bundle (Figure 1(b)) of a vector bundle (E, q, M) . First consider the horizontal dual. The canonical pairing of E ∗ with E prolongs to a pairing of T (E ∗ ) → T M with T E → T M . Suppose given X ∈ T (E ∗ ) and d d ξ ∈ T E with T (q)(X) = T (q∗ )(ξ ) . Then X = dt ϕt |0 ∈ T (E ∗ ) and ξ = dt et |0 ∈ T E , where et ∈ E and ϕt ∈ E ∗ can be taken so that q∗ (ϕt ) = q(et ) for t near zero. Now define the tangent pairing , by d ϕt , et . (22) X, ξ = dt 0 To show that this is nondegenerate it is sufficient to work locally. Suppose, therefore, that E = M ×V . Regard ξ as (x0 , v0 , w0 ) ∈ Tm0 M ×V ×V and X as (x0 , ϕ0 , ψ0 ) ∈ Tm0 M × V ∗ × V ∗ . Then d d X= (mt , ϕ0 + tψ0 ) , (mt , v0 + tw0 ) , ξ= dt dt 0 0 where

d dt mt |0

= x = T (q)(X) = T (q∗ )(ξ ) . So d X, ξ = ϕ0 + tψ0 , v0 + tw0 . dt 0

Expanding out the RHS, the constant term and the quadratic term vanish in the derivative, and we are left with X, ξ = ψ0 , v0 + ϕ0 , w0 from which it is clear that , is nondegenerate. We now need to establish that this is a pairing of the double vector bundles. Proposition 4.1. The tangent pairing , of T (E ∗ ) with T E over T M satisfies ∗, the conditions of Proposition 3.3. In particular, for m ∈ M and ϕ, ϕ1 , ϕ2 ∈ Em e, e1 , e2 ∈ Em , ϕ, e = 0, 0ϕ , e = ϕ, e,

0ϕ , 0e = 0, ϕ, 0e = ϕ, e

and τ∗ (ϕ1 , ϕ2 ), τ (e1 , e2 ) = ϕ1 , e2 + ϕ2 , e1 , where τ∗ and τ are the injections in the core sequences of T (E ∗ ) and T (E). Proof. These are easily verified from the definition. For example, ϕ = d e = dt (te)|0 , so

d dt (tϕ)|0

and


467

d 2 ϕ, e = t ϕ, e = 0, dt 0 whereas 0ϕ =

d dt ϕ|0 ,

so d tϕ, e = ϕ, e. 0ϕ , e = dt 0

The bilinearity conditions are easily verified and the final equation follows.

Thus the pairing of the cores of T (E ∗ ) and T (E) is the zero pairing, and so too is the pairing of the zero sections above E ∗ and E . However the core of T (E ∗ ) and the zero section of T (E) are paired under the standard pairing, and the same is true of the zero section of T (E ∗ ) and the core of T (E). It now follows that there is an isomorphism of double vector bundles from T (E ∗ ) to the dual T E × T M of T E over T M . For convenience we denote this simply by T • E and call it the prolongation dual of T E . The next result follows from the general theory of Section 3. Proposition 4.2 ([Mackenzie and Xu 1994]). The map I : T (E ∗ ) → T • (E) defined by I (X), ηT M = X, η, where X ∈ T (E ∗ ) , η ∈ T E , is an isomorphism of double vector bundles preserving the side bndles E ∗ and T M and the core bundles E ∗ . When a name is needed we call I the internalization map. In the future we will almost always work with T (E ∗ ) and the tangent pairing rather than with T • E and I . Now consider the vertical dual of T E . Since the core of the double vector bundle T E is E , dualizing the structure over E leads to a double vector bundle of the form rE T ∗E − −−→ E ∗ cE

⏐ ⏐ ? E

⏐ ⏐ ? qE ∗

(23)

−−−→ M. qE

We refer to this as the cotangent dual of T E . We will give a detailed description of the structures involved. Although this is a special case of the general construction, this example is so basic to the rest of the paper that it merits a specific treatment. In (23) the vertical bundle is the standard cotangent bundle of E , and the notation TX∗ (E) will always refer to the fibre with respect to cE . In this bundle we use standard notation, and denote the zero element of TX∗ (E) by 0∗X . We drop the subscripts E from the maps when no confusion is likely. The map r : T ∗ E → E ∗ takes the form

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K. C. H. Mackenzie

r(), Y = , τ (X, Y ) = , 0X + + Y , TX∗ (E) ,

where ∈ E ∗ we have

X ∈ Em and Y ∈ Em . Thus r() ∈

∗. Em

(24)

For the addition over

+∗ #, ξ + + η = , ξ + #, η, E

∗ , and ξ ∈ T (E) , where ∈ TX∗ (E) , # ∈ TY∗ (E) with r() = r(#) ∈ Em X ∗ η ∈ TY (E) with T (q)(ξ ) = T (q)(η) . This defines +∗ # ∈ TX+Y (E) . Similarly, E we have t E.∗ , t ξ = t, ξ ,

.

∗ , is 0rϕ ∈ for t ∈ R and ξ ∈ TX (E) . The zero element of r −1 (ϕ), where ϕ ∈ Em ∗ T0m (E) , where 0rϕ , T (0)(x) + X = ϕ, X

for x ∈ Tm (M), X ∈ Em . Given ω ∈ Tm∗ (M), the corresponding core element ω is ω, T (0)(x) + X = ω, x for x ∈ Tm (M), X ∈ Em . The injection over E , q ! T ∗ M → T ∗ E,

(X, ω) → 0∗X +∗ ω, E

is precisely the dual of T (q)! ; that is, it is the map corresponding to the lifting of 1-forms from M to E . Thus 0∗X E+∗ ω is the pullback of ω ∈ Tm∗ (M) to E at the point X ∈ Em . The core exact sequence for c is r ! =τ ∗ q ! T ∗ M >−−−> T ∗ E −−−2 q ! E ∗ ,

(25)

and this is the dual of the core exact sequence for T E and pE . The other core exact sequence is c! q∗! T ∗ M >−−−> T ∗ E −−−2 q∗! E, (26) where each bundle here is over E ∗ . The injection q∗! T ∗ M → T ∗ E is (ϕ, ω) → 0rϕ + ω and 0rϕ + ω, T (0)(x) + X = ϕ, X + ω, x. Given ω ∈ T ∗ M , the corresponding core element is ω = (ω, 0, 0). To summarize, the two dual double vector bundles of D = T E are D ×E = T ∗ E −→ E ∗ ⏐ ⏐ ?

⏐ ⏐ ?

E −→ M

D ×T M = T • E −→ T M and

⏐ ⏐ ?

⏐ ⏐ ?

E ∗ −→ M


469

and the pairing , f = , ξ E − f, ξ T M

(27)

for suitable ξ ∈ T E . Composing the isomorphism ZE from 3.4 with the dual over E ∗ of the internalization isomorphism I , we get an isomorphism of double vector bundles (I × E ∗ ) ◦ ZE : T ∗ E → T ∗ (E ∗ ); denote this temporarily by S −1 . For ∈ T ∗ E we have S −1 (), XE ∗ = (I ×E ∗ ) ◦ ZE (), XE ∗ = ZE (), I (X)E ∗ = , I (X) = , ξ E − I (X), ξ T M = , ξ E − X, ξ . Here we used the definition of ZE , the definition (27), and the definition of I . It follows that for F ∈ T ∗ (E ∗ ) , writing = S(F) , we have F, XE ∗ = S(F), ξ E − X, ξ . Recall that I , and hence its dual, preserves both sides and the core, whereas ZE induces − id on the sides E . We therefore define R : T ∗ (E ∗ ) → T ∗ (E),

R(F) = S( E−∗ F).

To summarize, we have the following. Theorem 4.3 ([Mackenzie and Xu 1994]). The map R just defined is an isomorphism of double vector bundles, preserving the side bundles E and E ∗ , and inducing − id : T ∗ M → T ∗ M on the cores. Further, for all ξ ∈ T E , X ∈ T (E ∗ ) , F ∈ T ∗ (E ∗ ) such that ξ and X have the same projection into T M , X and F have the same projection into E ∗ , and F and ξ have the same projection into E , X, ξ = R(F), ξ E + F, XE ∗ .

(28)

We call R the reversal isomorphism. It is proved in [Mackenzie and Xu 1994] that R is an antisymplectomorphism of the canonical symplectic structures.

5 Triple vector bundles The definition of a triple vector bundle follows the same pattern as in the double case. There are a number of evident reformulations. Definition 5.1. A triple vector bundle is a manifold III together with three vector bundle structures, over bases D1 , D2 , D3 , each of which is a double vector bundle with side bundles, respectively, E2 and E3 , E3 and E1 , E1 and E2 , where E1 , E2 , E3 are vector bundles over a shared base M , such that each pair of vector bundle structures on III forms a double vector bundle, the operations of which are vector bundle morphisms with respect to the third vector bundle structure.

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K. C. H. Mackenzie

We display a triple vector bundle in a diagram such as Figure 3(a). (We always read figures of this type with (III; D1 , D2 ; E3 ) at the rear and (D3 ; E2 , E1 ; M) coming out of the page toward the reader.) The three structures of double vector bundle on III are the upper double vector bundles, and D1 , D2 , D3 are the lower double vector bundles. We refer to (D1 ; E2 , E3 ; M) as the floor of III and to (III; D2 , D3 ; E1 ) as the roof of III . III −→ D2 ⏐ ⏐ ?

k 1 −→ d2 H⏐ H ⏐ H j HH j ⏐ ⏐H ? ? d3 −→ e1

H ⏐ H H⏐H j HH j

? D3 −→ E1

⏐ D1 −→ E3 ⏐ ?

H

HH j

H

HH j

⏐ ⏐ ?

d1 −→ e3

H

HH j

E2 −→ M (a)

⏐ ⏐ ?

H

HH j

⏐ ⏐ ?

e2 −→ m (b)

Fig. 3.

We have found that, rather than assembling a notation capable of handling any calculation in a triple vector bundle without ambiguity, it is generally preferable to develop an ad hoc notation for each occasion. The great majority of calculations use only certain parts of the structure, and in such cases a modification of the notation of Section 1 is often sufficient. Each of the lower double vector bundles Di has a core, which is denoted Ci . The core of the upper double vector bundle (III; D3 , D2 ; E1 ) is denoted K1 . Consider a 1 . Then the d in Figure 3(b) is core element k 1 ∈ III , where k1 projects to e1 ∈ Em 2 the zero over e1 for D2 → E1 , and d3 is the zero over e1 for D3 → E1 . From the morphism condition we then have that e2 and e3 are zeros over m . So d1 = c is a core element for some c ∈ C1 . This defines a map K1 → C1 . For k, k ∈ K1 over the same element of C1 , define k +C1 k = k +D1 k ,

(29)

where each of the three bars refers to the roof double vector bundle. With scalar multiplication defined in a similar fashion, K1 → C1 is a vector bundle and a double vector bundle as shown in Figure 4(a). The cores of the other upper double vector bundles are likewise denoted K2 and K3 and form double vector bundles as in Figure 4(b)(c). These three are the core double vector bundles. Although defined by restrictions of the operations in III , they are not substructures of III . Denote the core of (K1 ; C1 , E1 ; M) by W . In Figure 3(b), let k1 = w , where w ∈ W . Then c1 is the zero of C1 over m , and so d1 = c1 is a double zero of D1 .

Duality and triple structures K2 −→ E2

K1 −→ E1 ⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

471

K3 −→ E3

⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

C1 −→ M

C2 −→ M

C3 −→ M

(a)

(b)

(c)

Fig. 4. 3 Next, since e2 is a zero, (d3 ; e2 , e1 ; m) must be of the form d3 = 0D e1 +E2 c3 . But e1 is zero, since w is in the core, so d3 is a core element. But it is known to be a zero over e1 , so must be a double zero. Similarly, d2 is a double zero. This proves most of the next result, and the remainder is an easy verification.

Proposition 5.2. Each of the core double vector bundles has as core the set W of elements w ∈ III for which the projection to each of D1 , D2 , D3 is a double zero of the lower double vector bundle. Further, the vector bundle structures with base M induced on W by the various core double vector bundles coincide. Given w ∈ W , the core elements in III corresponding to w1 ∈ K1 , w 2 ∈ K2 , and w 3 ∈ K3 coincide. We call W the ultracore of III . Example 5.3. For a double vector bundle (D; A, B; M), the tangent prolongation triple vector bundle is as shown in Figure 5(a). Two of the three core double vector bundles are copies of (D; A, B; M) and the third is (T C; C, T M; M). The ultracore of T D is C , the core of D . It is illuminating to verify (29) and 5.2 directly in this example. T ∗ D −→ D × B

T D −→ T B

⏐ HH ⏐ HH j H j H ⏐ ⏐ ?

⏐ ⏐ ?

? T A −→ T M

⏐ D −→ B ⏐ ?

H

HH j

H

HH j

⏐ ⏐ ?

HH ⏐ j⏐ H

?D × A

D −→

H

⏐ B ⏐ ?

HH j

A −→ M (a)

H A

HH j

−→ M

(b) Fig. 5.

The key to understanding the relations between the duals of a double vector bundle and the role of the dihedral group (21) lies in constructing a cotangent form of this

472

K. C. H. Mackenzie

example. Both the left and the rear faces of Figure 5(a) are tangent prolongation double vector bundles of ordinary vector bundles and so we can form the figure in Figure 5(b). In Figure 6(a) we have added the two double vector bundle duals associated to D . In this diagram each of the four vertical sides, and of course the floor, is a double vector bundle. We need to prove that the roof is a double vector bundle and that Figure 6(a) is a triple vector bundle. First consider the roof, shown in Figure 6(b). We use a short notation for the projections. T ∗ D −→ D × B

rB T ∗ D −→ D × B

H H ⏐ HH⏐ HH ⏐ ⏐ j j H ? ?H

D × A −→ C ∗

D −→

B

⏐

⏐

A

−→ M

rA

⏐ H H⏐ ?H ? HH H j H j H

⏐ ⏐ ?

⏐ ⏐ ?

q×B

D × A −→ C ∗ q×A (b)

(a) Fig. 6.

In this structure, we know that each side is a vector bundle. Proposition 5.4. The structure in Figure 6(b) is a double vector bundle with core T ∗ C . Proof. First, we must prove that the projections form a commutative square. Take f ∈ Td∗ D , where d has the form (d; a, b; m) . Then, for all (d ; a, b ; m), 0d + +A d . rA (f), d = f, A

Here 0d is the zero of T D → D above d and the subscript on + +A indicates that this is the tangent of the addition in D → A . The superscript A on the bar indicates that D is here the core of (T D; T A, T M; A). Writing ϕ = rA (f) , we next have q ×A (ϕ), c = ϕ, 0D a +B c. Here 0D a is the zero of D → A over a and c is the core element of D corresponding to c . Writing out the corresponding formulas for the other side, we must prove that A

B

+B (0D +A c) . 0d + +A (0D a +B c) = 0d + b Using (29), the LHS becomes

(30)


473

A

+A (0D +B c). 0d + a + Writing in terms of tangents to curves, we have A d d d D D 0d = 0D = 0 ) = , d , (t 0 A a a dt 0 dt dt a 0 0

.

c=

d tc . dt 0

Now, using the interchange rule, D D d +A (0D a +B c) = (d +B 0b ) +A (0a +B c) D D = (d +A 0D a ) +B (0b +A c) = d +B (0b +A c)

and from this (30) follows. The proof that rA preserves the addition and scalar multiplication proceeds in a similar way. Next, we show that the core is T ∗ C . Suppose that f ∈ Td∗ D maps to zero under both rA and rB . Then d = c is a core element and f vanishes on elements ξ ∈ Tc D which are vertical with respect to either qAD or qBD . If ξ is vertical with respect to qAD then, in the notation of Figure 7(a), X = 0A m , and it follows that Z = 0m and D so Y is a core element. Likewise, if ξ is vertical with respect to qB , then Y = 0B m and X is a core element. Adding two such representative elements, it follows that f vanishes on all X, as shown in Figure 7(b).

ξ −→ Y

X −→ b

⏐ HH⏐ HH j H j H ⏐ ⏐ ?

⏐ HH ⏐ HH j H j H ⏐ ⏐ ? ? a −→ 0m

? X −→ Z

⏐ ⏐ c −→ 0B m ?

H

HH j

H

HH j

⏐ ⏐ ?

⏐ ⏐ c −→ 0B m ?

H

H

HH j

0A m −→ m (a)

HH j

⏐ ⏐ ?

0A m −→ m (b)

Fig. 7.

Now take ξ ∈ Tc D as shown in Figure 7(a). Because X ∈ T0Am A , it has the form X = T (0A )(Z) + a for some a ∈ Am ; likewise Y has the form Y = T (0B )(Z) + b for some b ∈ Bm . Now define X = (T (0D +A +B 0c ) + (T (0D 0c ). B )(b) + A )(a) + D

Then γ = ξ − X has the form shown in Figure 8(a) and is an element of T C . D

It is now possible to extend a given ω ∈ Tc∗ C to ω ∈ Tc∗ D by

474

K. C. H. Mackenzie

D×B

γ −→ T (0B )(Z)

⏐ HH ⏐ HH ⏐ H⏐ H H HH ? ?H j j c −→

H

0B m

T (0A )(Z) −→ Z

H ⏐ H⏐ ?H HH HH j j

HH

0A m

H

⏐ HH j ⏐ × ?D A −→ C ∗ D −→

⏐ ⏐ ?

H

⏐ B⏐ ?

HH j

−→ m

H

A

HH j

⏐ ⏐ ?

−→ M

(b)

(a) Fig. 8.

ω, ξ = ω, ξ − X D

and ω is annulled by both rA and rB . This ω is the core element of the double vector bundle in Figure 6(b). Now that the commutativity of the projections has been established, verification that addition and scalar multiplication are preserved is straightforward.

The double vector bundle in Figure 6(b) is of a type not previously encountered. It is now a straightforward matter to complete the proof of the following. Theorem 5.5. The structure in Figure 6(a) is a triple vector bundle. The core double vector bundles are (T ∗ A; A, A∗ ; M), (T ∗ B; B, B ∗ ; M) and and the ultracore is T ∗ M . Observe that the triple vector bundle ∗ T D has a much higher degree of symmetry than T D . (T ∗ C; C, C ∗ ; M),

Example 5.6. Consider seven vector bundles E1 , E2 , E3 , C1 , C2 , C3 , W over a shared base M . Let D1 be the trivial double vector bundle with sides E2 and E3 and core C1 , and likewise form D2 and D3 . Similarly, let K1 be the trivial double vector bundle with sides C1 and E1 and core W , and form K2 and K3 in the same way. Lastly, let III be the pullback of all seven vector bundles over M . Then III can be considered as the trivial double vector bundle with side bundles D1 → E3 and D2 → E3 and core K3 → E3 . Likewise, III can be considered the trivial double vector bundle over D2 and D3 with core K1 and over D3 and D1 with core K2 . With these structures, III is a triple vector bundle, the trivial triple vector bundle determined by the given seven vector bundles. More refined versions of this construction exist. For example, suppose given four vector bundles E1 , E2 , E3 , W on M and three double vector bundles (D1 ; E2 , E3 ; M), (D2 ; E3 , E1 ; M), (D3 ; E1 , E2 ; M). Then there is a triple vector bundle for which D1 , D2 , D3 are the lower double vector bundles and W is the ultracore, and for which each of the core double vector bundles is trivial.


475

6 Cornerings Continue with a double vector bundle D as in the previous section. Since D is a vector bundle over A , we have T ∗ D ∼ = T ∗ (D × A) by 4.3, and similarly ∗ ∗ × T D ∼ = T (D B) . Once it has been shown that these isomorphisms respect the triple structures, we can regard 3 as acting on the cube T ∗ D by rotations about the axis from T ∗ D to M . Theorem 6.1. The map R −1 : T ∗ D → T ∗ (D × A) arising from the vector bundle D → A is an isomorphism of triple vector bundles over ZB : D × B → (D × A × C ∗ ) , the other maps on the side structures being identities. Proof. The main work is to show that R −1 is a morphism of vector bundles over ZB . Take ∈ Td∗ D and denote R −1 () by f . Let d have the form (d; a, b, m) and let the projections of to D × A , D × B , and C ∗ be χ , ψ , and κ , respectively. Since R preserves D and D × A , it follows that f projects to d ∈ D and to χ ∈ D × A . For ψ we have, from (24), B ψ, d1 B = , 0d + + B d 1 D

(31)

for any d1 of the form (d1 ; a1 , b; m). For f and we have, by (28), X, ξ T A = , ξ D + f, XD × A ,

(32)

where X ∈ T (D × A) has the form (X; χ , X; a) for some X ∈ T A , and ξ ∈ T D then has the form (ξ ; d, X; a) . Next, for ZB (ψ) ∈ D × A × C ∗ , we have, for each ϕ ∈ D × A of the form (ϕ; a2 , κ; m) , ZB (ψ), ϕ = ϕ, ψ

C∗

= ϕ, d2 A − ψ, d2 B

(33)

for any d2 ∈ D of the form (d2 ; a2 , b; m). Lastly, for the same ϕ we have (D 0χ rC ∗ (f), ϕ = f,

× A)

+ +C ∗ ϕ (D

(D × A)

× A)

.

(34)

×

is the zero in T (D × A) over χ and ϕ (D A) is the core element of Here 0χ T (D × A) corresponding to ϕ . The addition is in the bundle T (D × A) → T C ∗ . We must prove that the RHSs of (33) and (34) are equal. We substitute (D X = 0χ

× A)

+ +C ∗ ϕ (D

× A)

and

ξ = 0d + +B d 1

B

into (32). Providing a1 = a2 , the relevant projections match. Now applying (iv) of Proposition 3.3 to the double vector bundles (T (D × A); T A, T C ∗ ; T M) and (T D; T A, T B; T M), we have (D × A)

0χ X, ξ T A =

(D × A)

= 0χ

+ +C ∗ ϕ (D

× A)

, 0d + +B d 1 T A

, 0d T A + ϕ (D

B

× A)

B

, d 1 T A .

476

K. C. H. Mackenzie (D × A)

In the first term, 0χ

is tangent to the path constant at χ , and 0d is tangent to ×

(D A) , 0d T A is tangent to the path constant at the path constant at d ; therefore, 0χ × χ , dA , and is therefore zero. For the second term, ϕ (D A) is tangent to the path × B B t C.∗ ϕ and d 1 is tangent to the path t B. d1 , so ϕ (D A) , d 1 T A is tangent to the path t C.∗ ϕ, t B. d1 A and by (v) of Proposition 3.3 this is tϕ, d1 A . Altogether, we have that X, ξ T A = ϕ, d1 A . Using (31), we have that the RHS of (34) is

ϕ, d1 A − ψ, d1 B and this is equal to the RHS of (33) by the proof of 3.2. The rest of the proof is now straightforward.

For a single vector bundle E → M , the pairing of E ∗ with its dual E ∗∗ can be identified in a straightforward way with the pairing of E with its dual. For double vector bundles it is first necessary to ensure that pairings are chosen in a consistent way. Consider a double vector bundle (D; A, B; M) and assign signs to the two upper structures as in Figure 9(a) in order to show that we pair the duals according to (17). Now, referring to Figure 8(b), we assign signs in such a way that each of A, B, C ∗ has one positive and one negative arrow approaching it, and each of D , D × A , D × B has one positive and one negative arrow departing from it; see Figure 9(b)(c). We therefore, for example, take the pairing of the duals of D × A to be D, D × A × C ∗

B

= D × A, D × A × C ∗ C ∗ − D, D × AA .

⏐ ⏐ ⊕ ?

⊕ D × B −→ B

⊕ D × A −→ C ∗

3 D −−−→ B ⏐ ⏐ ?

3

A −−−→ M

⏐ ⏐ ?

⏐ ⏐ ?

A

−→ M

(a)

3

⏐ ⏐ ?

⏐ ⏐ ?

C ∗ −→ M (c)

(b)

Fig. 9.

Proposition 6.2. For the isomorphism ZB : D × B → (D × A × C ∗ ) , , #

C∗

= , ZB (#)C ∗ ,

(35)

d, #B = − d, ZB (#)

for compatible ∈ D × A , # ∈ D × B , d ∈ D .

B


477

Proof. The first is the definition of ZB . The second follows from ZB × C ∗ = ZA . If we insert these equations into (35), we get (17). Thus the signing on D × A is compatible with that on D . For ordinary vector bundles E1 and E2 on the same base M , one could take the view that a pairing of E1 with E2 is what enables one to construct a cotangent double vector bundle with sides E1 and E2 . In a similar way, three double vector bundles with suitably overlapping sides can be completed to a cotangent triple vector bundle if and only if any two of them are the duals of the third. Definition 6.3. Consider three double vector bundles as in Figure 10(a), together with six pairings: , E1 of D2 and D3 over E1 , , E2 of D3 and D1 over E2 , , E3 of D1 and D2 over E3 , and , 1 of C1 and E1 over M , , 2 of C2 and E2 over M , , 3 of C3 and E3 over M , such that each pairing of D bundles is a pairing of double vector bundles ( as defined in Proposition 3.3 ) with respect to the pairing of the relevant cores and sides. Then if D2 , D3 E1 = D1 , D2 E3 − D1 , D3 E2 holds, we say that the system is a cornering of D1 with D2 and D3 .

T (T ∗ E) −→ T (E ∗ )

D3

⏐ HH j H ⏐ ? D2 −→ E1

⏐ D1 −→ E2 ⏐ ?

H

H Hj HH H j

⏐ HH ⏐ HH ?

⏐HH ⏐ HH ?

H j H

⏐ ⏐ ?

TE

⏐ H ⏐ ⏐ HH H⏐ ?H ? HH HH j H j H

H

E3 −→ M

−→ T M

H j H

T ∗ E −→ E ∗

E −→ M

(a)

(b) Fig. 10.

Clearly, choosing any double vector bundle in a cornering, the other two double bundles may be identified with its duals and the cornering may be identified with the lower sides of the cotangent triple vector bundle associated with the chosen double. Remark 6.4. For an ordinary vector bundle E one may form the cotangent triple of D = T E . Now the canonical diffeomorphism between T ∗ T E and T T ∗ E [Abraham and Marsden 1985] is, since E is a vector bundle, an isomorphism of double vector bundles, and so the triple T ∗ T E is isomorphic to the tangent prolongation of T ∗ E , as shown in Figure 10(b). Now the pairing of the bundles over E in the left face gives rise to the canonical 1-form on T ∗ E , and the pairing of the bundles in the roof gives rise to the canonical 1-form on T ∗ E ∗ .

478

K. C. H. Mackenzie

7 Duals of triple vector bundles Consider now a general triple vector bundle III as in Figure 3(a). Dualize III over the base D1 . Each of the upper double vector bundles of which III → D1 is a side has a dual which is familiar from Section 4. Following the example of 5.5, we complete the cube as in Figure 11(a). III× D1 −→ K3 × E3

IIIPY −→ D1

H H ⏐ HH ⏐ HH ⏐ ⏐ H?H HH ? j j

D1

−→

H

E3

⏐ ⏐ ?

K2 × E2 −→ W ∗

⏐ H ⏐ ⏐ H⏐ ?H ? HH HH j j

HH

E2

−→ M

(a)

H

H HH⏐ HH ⏐ HH ?HH j j

D2 −→ E3

D3P −→ E2

⏐ H H ⏐ ⏐ ⏐ HH H ?H ? HH HH j j E1 −→ M (b)

Fig. 11.

Theorem 7.1. There is a triple vector bundle as shown in Figure 11(a) in which the four vertical sides are dual double vector bundles as just described. We omit the details of this. As with the case III = T D , five of the six faces are double vector bundles of known types and the main work is to show that the roof— which belongs to a new class of examples—is a double vector bundle, and calculate its core, which is K1 × C1 . The proof follows exactly the same outline as in 5.4, though steps involving derivatives must be replaced with forms of the interchange laws. Notice that in Figure 11(a), two of the three upper double vector bundles are standard duals of the double vector bundles in the corresponding positions in Figure 3(a). Two of the lower double vector bundles are duals of core double vector bundles of III . The core double vector bundles of III × D1 are given in Figure 12. The ultracore is E1∗ , the dual of the bundle which in the original was diagonally opposite III in the plane perpendicular to the axis of dualization. The relationship between the three duals of III is embodied in the cotangent quaternary vector bundle of III , as shown in Figure 13. Denote dualization of III along the three axes by X , Y , and Z . In terms of Figure 3(a), take Z to be dualization along the vertical axis, Y to be along D3 and X to be along D2 . Compositions such as ZXZ are triple versions of the operation P studied in Section 3. Precisely, applying ZXZ to III in Figure 3(a) applies P to the rear face and to the front face; denote this by PY . This operation may also be regarded as reflection of III in the plane through III , D3 , M , and E3 ; see Figure 11(b). Notice that each face has been flipped in the sense that it cannot be returned to its original position by a proper rotation of the cube. Further, the core double vector bundle which


479

lies in the plane through III , D3 , M , and E3 is left fixed; the other two are flipped and interchanged. With similar definitions of PX and PZ , we have PX = Y ZY = ZY Z,

PY = ZXZ = XZX,

PZ = XY X = Y XY,

(36)

each of PX , PY , PZ having order 2. Equivalently, each of XY , Y Z , ZX has order 3. New in the triple case are the products QZ = ZXY Z , QX = XY ZX and QY = Y ZXY and their inverses. It is easily found from (36) that QX , QY , and QZ have order 3 and that QZ QY QX = I . Curiously, the equation QX QY QZ = I or, equivalently, (XY Z)4 = I , is not a consequence of (36), but it may be verified directly by calculating the effect on III . We now have: Theorem 7.2. The group of operations on III generated by X , Y , and Z satisfies the relations X2 = I , Y 2 = I , Z 2 = I , (XY Z)4 = I , (Y ZX)4 = I , (ZXY )4 = I , together with (36). By a calculation with [GAP], the group defined by these relations has order 72. Denote the group of operations generated by X , Y , and Z by VB3 . It is straightforward to find more than 36 distinct elements of VB3 and so it must have order 72. It thus cannot be, as one might have expected, a subgroup of the full symmetry group of the hypercube, which has order 384 [Coxeter 1973]. This shows that the situation with double vector bundles, in which the operations generated by dualization can be identified with symmetries of the cotangent triple, does not extend in the analogous fashion to triple vector bundles and symmetries of the hypercube.

8 General principles On the basis of the duality theory for duals and triples, we may formulate some likely principles for the duality of general multiple vector bundles. It may be that the proofs are mainly a matter of acquiring sufficient motivation and notation, but we cannot rule out the possibility that new phenomena arise with increasing dimension. There are three groups associated with an n -fold vector bundle N . First, the various operations generated by flips of the constituent double vector bundles generate an K1 × C1 −→ W ∗

D2 × E3 −→ C2∗

D3 × E2 −→ C3∗

⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

⏐ ⏐ ?

C1

−→ M

E3

−→ M

E2

−→ M

(a)

(b) Fig. 12.

(c)

480

K. C. H. Mackenzie

T ∗ III −→ III× D2 ⏐ @ ⏐ ? @

⏐ ⏐ ?

@

@

@

×E III× D1 −→ K3@ 3

III −→ D2

⏐ @ ⏐@ ⏐ @⏐ ? ? @

@

@ @ @ @ @ @ @ @ @ @ @ @ @ @ @ @ @ R @ R @ @ @ × D −→ K × E III@ @ 3 1 1 @ ⏐@ ⏐ ⏐ @ ⏐ @ ? ? @ @ @ @ R× @ R ∗ @

@ @ @ D1 −→ E3 @ @ @ @ @ @ @ @ @ @ @ @ @ @ @ @ R @ @ R @ @ @ @ D3 −→ E1 @ @ ⏐ ⏐ ⏐ @ @⏐ ? ? @ @ @ @ R @ R @

@

K2 E2 −→

W

E2 −→ M Fig. 13.

action of the symmetric group Sn . Secondly, there is an obvious sense in which individual n -fold vector bundles may have more symmetry than others, as we remarked in the case of T ∗ D and T D in Section 5. Of most interest, however, is the group VBn generated by the dualization operations. We have seen that VB2 is S3 and that VB3 has order 72. Further, the subgroup of VB3 generated by XY XZ , Y ZY X , and ZXZY has order 12 and is normal, with quotient isomorphic to S3 . In the general case, the n duals of an n-fold vector bundle N and N itself form the (n + 1) lower n -faces of an (n + 1) -fold vector bundle, which may be completed to be the cotangent (n + 1) -fold vector bundle of N , or of any of the duals of N . The (n + 1) upper n -faces of T ∗ N consist of the n cotangent n-fold vector bundles of the upper (n − 1) -faces of N , together with one n -fold vector bundle of a new type, which incorporates data from all of the structure of N . It is reasonable to conjecture that if X1 , . . . , Xn denote the dualization operations, each of order 2, then we have, for each 1 k n and each string i1 , i2 , . . . , ik of k distinct elements of {1, . . . , n} ,


481

(Xi1 Xi2 · · · Xik )k+1 = 1. Note added in proof It has been pointed out to me by Alfonso Gracia-Saz that the calculation in Theorem 7.2 is incomplete. A complete account will be provided in a subsequent article. Acknowledgments I am grateful to Moty Katzman for introducing me to the GAP software, which was very valuable in Section 7.

References R. Abraham and J. Marsden, Foundations of Mechanics, 2nd ed., Addison–Wesley, Reading, MA, 1985. A. Coste, P. Dazord, and A. Weinstein, Groupoïdes symplectiques, in Publications du Département de Mathématiques de l’Université de Lyon, I, number 2/A-1987, Département de Mathématiques, Université de Lyon, Lyon, 1987, 1–65. T. J. Courant, Dirac manifolds, Trans. Amer. Math. Soc., 319 (1990), 631–661. H. S. M. Coxeter, Regular polytopes, Dover, New York, 1973. GAP, GAP: Groups, Algorithms, and Programming, Version 4.3, The GAP Group, St. Andrews, Fife, UK, 2002; www.gap-system.org. K. Konieczna and P. Urban´ ski, Double vector bundles and duality, Arch. Math. ( Brno ) , 35-1 (1999), 59–95. J.-H. Lu and A. Weinstein, Groupoïdes symplectiques doubles des groupes de LiePoisson, C. R. Acad. Sci. Paris Sér. I Math., 309 (1989), 951–954. K. C. H. Mackenzie, On symplectic double groupoids and the duality of Poisson groupoids, Internat. J. Math., 10 (1999), 435–456. K. C. H. Mackenzie, On certain canonical diffeomorphisms in symplectic and Poisson geometry, in Quantization, Poisson Brackets and Beyond ( Manchester, 2001) , Contemporary Mathematics, Vol. 315, American Mathematical Society, Providence, RI, pages 187–198. K. C. H. Mackenzie, General Theory of Lie Groupoids and Lie Algebroids, Cambridge University Press, Cambridge, UK, 2004. K. C. H. Mackenzie and P. Xu, Lie bialgebroids and Poisson groupoids, Duke Math. J., 73-2 (1994), 415–452. J. Pradines, Fibrés vectoriels doubles et calcul des jets non holonomes, Esquisses Mathématiques 29, Université d’Amiens, U.E.R. de Mathématiques, Amiens, France, 1974. J. Pradines, Remarque sur le groupoïde cotangent de Weinstein–Dazord, C. R. Acad. Sci. Paris Sér. I Math., 306-13 (1988), 557–560. A. Weinstein, Symplectic groupoids and Poisson manifolds, Bull. Amer. Math. Soc. ( N.S.) , 16 (1987), 101–104. A. Weinstein, Coisotropic calculus and Poisson groupoids, J. Math. Soc. Japan, 40 (1988), 705–727.

Star exponential functions as two-valued elements∗ Y. Maeda1 , N. Miyazaki2 , H. Omori3 , and A. Yoshioka4 1 Department of Mathematics

Faculty of Science and Technology Keio University Hiyoshi, Yokohama, 223-8522 Japan [email protected] 2 Department of Mathematics Faculty of Economics Keio University Hiyoshi, Yokohama, 223-8521 Japan [email protected] 3 Department of Mathematics Faculty of Science and Technology Tokyo University of Science Noda, Chiba, 278-8510 Japan [email protected] 4 Department of Mathematics Faculty of Science Tokyo University of Science Kagurazaka, Tokyo, 102-8601 Japan [email protected] Abstract. We propose a relatively new notion of two-valued elements, which arise naturally in constructing star exponential functions of the quadratics in the Weyl algebra over the complex number. This notion enables us to describe group-like objects of the set of star exponential functions of quadratics in the Weyl algebra.

1 Introduction Classically, geometries are described within the framework of manifolds which are distinguished among the topological spaces. The question may arise if there are ge∗ This research was partially supported by Grants-in-Aid for Scientific Research 15204005

(first author), 15740045 (second author), 14540092 (third author), and 15540094 (fourth author) from the Ministry of Education, Culture, Sports, Science, and Technology of Japan.

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ometries. In this paper, we attempt to propose a notion of two-valued elements, which seems to renew a geometric concept. A nontrivial example of objects we propose in this paper is given by the HopfH S1 fibering S 3 → S 2 . Viewing S 3 = q∈S 2 Sq1 (disjoint union), we consider the double H covering S˜q1 of each fiber S˜q1 , and the disjoint union q∈S 2 S˜q1 which is denoted by S˜ 3 . When S˜ 3 is considered as a point set, we are able to define local trivializations of S˜ 3 |Vi ∼ = Vi × S˜ 1 naturally through the trivializations S 3 |Vi given on a simple open covering {Vi }i∈ of S 2 . This structure permits us to treat S˜ 3 as a local Lie group, and hence itHlooks like a topological H space. On the other hand, we have a projection π : S˜ 3 = q∈S 2 S˜q1 → S 3 = q∈S 2 Sq1 as the union of fiberwise projections, as if it were a nontrivial double covering. S˜ 3 cannot be a manifold, since S 3 is simply connected. This might suggest us to make the notion of points vague. In particular, the “points’’ of S˜ 3 should be regarded as two-valued elements with ± ambiguity. We now consider a one-parameter subgroup S 1 of S 3 and the inverse image −1 S 3 are “two-valued", this simply can be considered both π (S 1 ). Since all points of 1 on S × Z2 and the double covering group, i.e., in some restricted region, this object can be regarded as a point set in several ways. In such a region, the ambiguity only arises if these two pictures of point sets are confused. Similar phenomena appear in constructing star exponential functions of quadratic forms in the suitably extended Weyl system, which leads us to explore a new type of geometry with a noncommutative (quantum) aspect. In [9], we have exhibited strange phenomena which violate the associativity for the Weyl algebra over C generated by two generators u and v. Furthermore, we have shown that the Lie algebra over C of quadratic forms can be exponentiated to a “group’’ which acts like a double covering group of simply connected group SLC (2), or the complexification of the metaplectic group Mp(2, R). As a sequel to [9], we continue these resutls to the case of Weyl algebra with 2m-generators u1 , . . . , um , v1 , . . . , vm , and show that similar phenomena occur. We show that star exponential functions can be viewed as two-valued elements. We note that an approach using gerbes may also describe such phenomena (see [3, 4, 9]), which would also give rise to a new geometrical formulation.

2 Weyl algebra and orderings 2.1 Weyl algebra The Weyl algebra W is the algebra over C generated by u1 , . . . , um , v1 , . . . , vm with the following commutation relations: [ui , vj ] = −iδij ,

(1)

where is a positive constant and [a, b] = a ∗ b − b ∗ a. Here the product on W is denoted by ∗. For abbreviation, we set u = (u1 , . . . , um ), and z = (u, v) =

Star exponential functions as two-valued elements

485

(u1 , . . . , um , v1 , . . . , vm ). Let Sym(2m, C) be the set of complex symmetric matrices A = (Aij ). For A ∈ Sym(2m, C), we define a quadratic form by A∗ (z) =

2m i,j =1

1 Aij (zi ∗ zj + zj ∗ zi ). 2

(2)

Denote by A the set of A∗ (z), where A ∈ Sym(2m, C). It is easily seen that A forms a complex Lie algebra isomorphic to spC (m). 2.2 Orderings Orderings are treated in the physical literature (see [1]) of quantum mechanics as the rule of association from c-number functions to q-number functions. There are typical orderings, called the standard ordering, the antistandard ordering and the Weyl ordering, and the in case of complex variables ζk = uk + ivk , ζl∗ = ul −ivl , the normal ordering, the antinormal ordering, and the Weyl ordering. However, from the mathematical view point, it is better to go back to the original understanding of Weyl which says that the ordering is the problem of realization of the Weyl algebra W . Since the Weyl algebra is the universal enveloping algebra of a Heisenberg Lie algebra, the Poincaré–Birkhoff–Witt theorem shows that this algebra can be viewed as an algebra defined on the space of polynomials. For precise formulations of ordering prescriptions in formal deformation quantization, one can refer to the article [2], but the theory using a formal deformation parameter is only a probe for genuine quantum theory. We emphasize here that the deformation parameter in this note is not a formal parameter, but a parameter in the positive reals. Thus we generalize orderings as follows. Let J be a 2m × 2m matrix defined by J = [ I0m −I0m ]. For every symmetric complex 2m × 2m matrix K = (K ij ), we set the product ⎧ ⎛ ⎞⎫ 2m ⎨ i ⎬ ← − − → ⎝ f (z) ∗K g(z) = f exp (3) ∂zi ij ∂zj ⎠ g, ⎩2 ⎭ i,j =1

where = ( ij ) = (K ij + J ij ). The product formula (3) is well defined for all f, g ∈ C[z], where C[z] = C[z1 , . . . , z2m ], and this satisfies zi ∗K zj − zj ∗K zi (= [zi , zj ]∗K ) = iJ ij ,

(4)

giving the same commutation relations (1) as the Weyl algebra W . Proposition 2.1. For every complex symmetric 2m × 2m matrix K, (C[z], ∗K ) forms an associative algebra isomorphic to W . Proposition 2.1 gives a realization of the Weyl algebra W , and at the same time it also gives a way to compute expressions in the Weyl algebra W . For instance, computing ui ∗ uj ∗ uk by (3) gives an expression of ui ∗ uj ∗ uk as a polynomial.

486


Thus the product formula (3) will be referred to as K-ordering, i.e., giving an ordering is necessary to a product formula which gives the Weyl algebra W once the generators are fixed. Note that according to the choice of K: 5 4 5 4 5 4 0 −Im 00 0 Im , , , Im 0 −Im 0 00 the product formulas (3) gives the standard ordering, the antistandard ordering and the Weyl ordering, respectively. By these formulation of orderings, intertwiners between K-orderings are explicitly given as follows. Proposition 2.2. For every pair of complex symmetric 2m × 2m matrices K, K , we have the intertwiner T : (C[z], ∗K ) → (C[z], ∗K ) defined as ⎞ ⎛ (5) (K ij − K ij )∂zi ∂zj ⎠ f. T (f ) = exp ⎝ 2i i,j

Namely, the identity T (f ∗K g) = T (f ) ∗K T (g),

(6)

holds for any f, g ∈ C[z]. With the precise statement given in a forthcoming paper, the intertwiner can be extended to a certain class of functions. However, as has been shown in [9] the intertwiner behaves only as a 2-to-2 mapping in the space of exponential functions of quadratic forms, since a square root appears in the amplitude part of intertwined functions. We think this is a basic phenomena which breaks the associativity of the ∗-product on the closed linear hull of the exponential functions of quadratic forms. Such strange phenomena occur only in the case that the deformation parameter is a nonformal parameter. In spite of this, it is important that one can consider one-parameter subgroups via the theory of ordinary differential equations.

3 Star exponential functions 3.1 Star exponential functions tA (z)

We give the explicit formula for the star exponential function e∗ ∗ for a fixed Kordering. For A ∈ Sym(2m, C), we denote by A[z] the symmetric quadratic function defined by 2m A[z] = Aij zi zj . (7) i,j =1

Set C× = C − {0}, and denote by F the set defined by


F = {F = g exp Q[z] | g ∈ C× , Q ∈ Sym(2m, C)}.

487

(8)

For A ∈ Sym(2m, C), we set A∗K (z) =

2m i,j =1

1 Aij (zi ∗K zj + zj ∗K zi ). 2

(9)

The product formula (3) gives A∗K (z) = A[z] + i Tr KA.

(10)

We realize the star exponential function of A∗K (z), for A ∈ Sym(2m, C) with the tA∗K (z)

help of the K-ordering. Namely, in order to get the formula for e∗K FK (t) =

tA∗ (z) e∗K K ,

and consider the following equation: + ∂t FK (t) = A∗K (z) ∗K FK (t), FK (0) = 1.

, we set

(11)

By the product formulas (3) and (9), the evolution equation (11) can be expressed as a differential equation. Thus the real analytic solution is unique, if it exists. By setting FK (t) = gK (t) exp QK (t)[z],

where QK (t) ∈ Sym(2m, C),

(12)

the evolution equation (11) is reduced to a system of ordinary differential equations on gK (t) and QK (t)[z]. By a direct, although rather complicate computation, we have the following. Theorem 3.1. The evolution equation (11) has a unique analytic solution FK (t) ∈ F explicitly given by FK (t) = gK (t) exp QK (t)[z], (13) where J QK (t) = − (tan tJ A) · (I − iK tan tJ A)−1 , gK (t) = (det(cos tJ A − iK sin tJ A))−1/2 .

(14) (15)

Remark. Maillard [5] also obtained this product formula by solving the successive power series of a Riccati-type equation. Note also that for every t ∈ C there is K-ordering such that FK (t) is well defined. The formula (13) for the star exponential functions of A∗K (z) specializes to the standard ordering and the Weyl ordering by plugging in K = [ I0m Im0 ] and K = 0, respectively. In particular, we have the following.

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Y. Maeda, N. Miyazaki, H. Omori, and A. Yoshioka tA∗ (z)

Corollary 3.2. For any A ∈ Sym(2m, C), the star exponential function e∗ expressed as −J e∗tA∗ (z) = det(cos tJ A)−1/2 · exp (tan tJ A)[z]

is

(16)

via the Weyl ordering. 3.2 Star exponential functions of rank one quadratics We examine the equation (11) for rank one quadratics. m For x = (x1 , . . . , xm ) and y = (y x, y = m 1 , . . . , ym ) ∈ C , we set i=1 xi yi . m m For a, b ∈ Cm , we consider a, u = i=1 ai ui and b, v = i=1 bi vi as elements of W . It is easy to see that [a, u, b, v]∗ = −ia, b.

(17)

Hence, if a, a = 1, then a, u and a, v form a canonical conjugate pair. Let m−1 m−1 SC = {a ∈ Cm | a, a = 1}. For every a ∈ SC , and α, β, γ ∈ C, we consider a quadratic form B∗ (α, β, γ ) = αa, u ∗ a, u + βa, v ∗ a, v + γ (a, u ∗ a, v + a, v ∗ a, u),

(18)

which is called a rank one quadratic form. In the following, we assume that the discriminant D = γ 2 − αβ = 1. We now write down the star exponential for the rank one quadratic form B∗ (α, β, γ ). We denote by FM (α, β, γ ) and FN (α, β, γ ) the solution of (11) for A∗ (z) = B∗ (α, β, γ ) with respect to K = 0 and [ I0m Im0 ], respectively. Then we have the following (see also [9]). m−1 Corollary 3.3. Assume that D = γ 2 − αβ = 1. Then for a ∈ SC , we have

FM (t, α, β, γ ) = gM (t, α, β, γ ) · exp QM (t, α, β, γ ),

(19)

where gM (t, α, β, γ ) = (cos t)−1 , 1 QM (t, α, β, γ ) = (tan t) · (αa, u2 + βa, v2 + 2γ a, ua, v).

(20) (21)

Similarly, we have FN (t, α, β, γ ) = gN (t, α, β, γ ) · exp QN (t, α, β, γ ).

(22)

Here gN and QN are given by gN (t, α, β, γ ) = e−i tγ · (cos 2t − iγ sin 2t)−1/2 ,

(23)


QN (t, α, β, γ ) =

1 (XN (t)a, u2 + YN (t)a, v2 + 2ZN (t)a, u ◦ a, v), ⎧

α sin 2t ⎪ X (t) = ⎪ N ⎪ 2 cos 2t−iγ sin 2t , ⎨ β 2t YN (t) = 2 cos 2sin t−iγ sin 2t ,

⎪ ⎪ ⎪ 1 ⎩ZN (t) = i 1 − 2 cos 2t−iγ sin 2t

where

489

(24)

(25)

and the ◦ in the product denotes the standard ordering.

4 Polar elements are two-valued elements 4.1 Polar elements Using the formulas of the star exponential functions (19) and (22), we show how two-valued elements appear. An idea of justifications of the star exponential function of quadratic forms B∗ (α, β, γ ) is to consider the star exponential functions expressed by the standard ordering and the Weyl ordering. Looking at the formulas in Corollary 3.3 and evaluating at t = 2π , we have that FM ( 2π , α, β, γ ) diverges, while FN ( 2π , α, β, γ ) is finite. Thus we think of FN ( 2π , α, β, γ ) as a realization of the star exponential function π of 2 B∗ (α, β, γ ), which is denoted by exp∗ ( 2π B∗ (α, β, γ )). However, by the formula (22) in Corollary 3.3, we obtain the following. m−1 Theorem 4.1. Assume a ∈ SC . For any (α, β, γ ) with γ 2 − αβ = 1, we have

exp∗

π 2

√ 2i a,u◦a,v B∗ (α, β, γ ) = −1e◦ ,

(26)

which is independent of the choice of α, β, γ . √ We will show that the ambiguity of −1 cannot be eliminated for all (α, β, γ ). m−1 . Definition 4.2. Assume a ∈ SC

ε00 (a) = exp∗

π 2

B∗ (0, 0, 1)

(27)

is called the polar element. 4.2 Two-valued elements m−1 We explain below that the polar elements ε00 (a), a ∈ SC act like two-valued elements. Since (α, β, γ ) = (0, 0, 1) and (0, 0, −1) are arcwise connected in the set

490


γ 2 − αβ = 1, and thus they have to be viewed as a single element. By Theorem 4.1, we have π

e∗2

(a,v∗a,u+a,u∗a,v)

=

2i √ a,u◦a,v −1e◦ π − 2 (a,v∗a,u+a,u∗a,v)

= e∗

(28) .

However, considering the exponential law of the ∗-exponential function t

e∗2


for t ∈ C − {singular set}, we must set π

e∗2


− π (a,v∗a,u+a,u∗a,v) e∗ 2

2i

= ie◦

a,u◦a,v

,

2i a,u◦a,v

= −ie◦

(29) .

If one attempts to fix the sign ambiguity, the exponential law and (28) give π


∗ e∗2

π


∗ e∗

−1 = e∗2 = e∗2

π


π − 2 (a,v∗a,u+a,u∗a,v)

(30)

= 1.

We choose a continuous path of (α, β, γ ) from (0, 0, 1) to (0, 0, −1) for the case m = 1 concretely as follows: Set a, u = u, a, v = v and ε00 = ε00 (a). By a careful calculation, we see iθ

Ad(e∗2

(u2 +v 2 )

)e∗2tuv 2 −v 2 )+cos 2θ

= e∗t (sin 2θ (u

(31) 2uv)

.

Since the discriminant of the quadratic form of the right-hand side is identically 1, the πi

(u2 +v 2 )

π

uv

right-hand side is identically ε00 for t = 2π . In particular, Ad(e∗4 )e∗ = ε00 . iθ 2 +v 2 ) (u However, consider, for each θ, the one parameter subgroup Ad(e∗2 )e∗2tuv with π respect to t, t ∈ [0, 2 ]. • ε00 2θ

This line is identically ε00 .

1• −ε00 •

?

Star exponential functions as two-valued elements πi

We easily see that Ad(e∗4

(u2 +v 2 ) πi

Ad(e∗4

491

)e∗2tuv = e∗−2tuv . In particular,

(u2 +v 2 )

)ε00 = −ε00

by the exponential law. Move 2θ from 0 to π. Note also that by (31), (23), there is a singularity at 2θ = π2 , t = 4π . We also have in the standard ordering for D = 1, π

e∗2

(αa,u2 +βa,v2 +γ (a,u∗a,v+a,v∗a,u)

=

2i √ a,u◦a,v −1e◦ .

By the exponential law, we see that ε00 (a) satisfies −1 (a))2 = −1, ε00 (a)2 = (ε00

−1 ε00 (a) ∗ ε00 (a) = 1.

(32)

Therefore, we must conclude that the sign ambiguity cannot be eliminated. One 2i √ a,u◦a,v with the sign ambiguity. Similar phenomena has to set ε00 (a) = −1e◦ have been discussed by Olver [6]. By the above observation, the polar element ε00 (a) should be regarded as a twovalued element. Otherwise we obtain a contradiction 1 = −1. Only in this way can one permit the identity −ε00 (a) = ε00 (a). Since such a notion does not exist in the set theory, it is impossible to define ε00 (a) as a point in a point set. In what follows, we set π

ε00 (k) = e∗2

(uk ∗vk +vk ∗uk )

=

2i √ uk ◦vk −1e◦ ,

k = 1, 2, . . . , m.

These are all regarded as two-valued elements. Although it is natural to write ε00 (k) ∗ ε00 (l) = ε00 (l) ∗ ε00 (k), we simultaneously have the equality ε00 (k) ∗ ε00 (l) = −ε00 (l) ∗ ε00 (k)

(k = l).

Hence we have ε00 (k) ∗ ε00 (k) = ±1, but we see that ε00 (k)2 = −1. This is just the same as {±1}{±1} = {±1}, but {±1}2 = 1. Hence ε00 (k)2 behaves like an ordinary number in the extended Weyl algebra. In spite of this, ε00 (k) does not behave like an ordinary number i, since it is easy to see with the bumping identity (see [9]) that Ad(ε00 (k))uk = −uk ,

Ad(ε00 (k))vk = −vk .

Using this we easily have Ad(ε00 (1))

' m i=1

* bi ui

= −b1 u1 +

m

b i ui .

(33)

i=2

m−1 Since every a, u, a ∈ SC is translated to u1 by a symplectic transformation, we have in general the reflection w.r.t. a:

492


Ad(ε00 (a))b, u = b − 2a, ba, u, Ad(ε00 (a))b, v = b − 2a, ba, v

(34)

We introduce a notion called a blurred double covering group, which is a grouplike object formed by 2-valued elements [9]. Theorem 4.3. Ad(ε00 (a) ∗ ε00 (b)) generate SO(m, C), hence {ε00 (a) ∗ ε00 (b)} generate a blurred double covering group of SO(m, C). However, this blurred double cover has a point set picture as SO(m, C) × C× . If a, b are restricted to real vectors, then Ad(ε00 (a)∗ε00 (b)) generate SO(m), hence {ε00 (a)∗ε00 (b)} generate a blurred double covering group of SO(m), which may be viewed as Spin(m).

References [1] G. S. Agawal and E. Wolf, Calculus for functions of noncommuting operators and general phase-space method of functions, Phys. Rev. D, 2-10 (1970), 2161–2186. [2] M. Bordemann, N. Neumaier, M. Pflaum, and S. Waldmann, On representation of star product algebra over cotangent spaces on Hermitian line bundles, J. Functional Anal., 199 (2003), 1–47. [3] J. L. Brylinski, Loop Spaces, Characteristic Classes and Geometric Quantization, Progress in Mathematics, Vol. 107, Birkhäuser, Boston, 1993. [4] N. Hitchin, Lectures on special Lagrangian submanifolds, in C. Vafa and S.-T. Yau, eds., Winter School on Mirror Symmetry, Vector Bundles and Lagrangian Submanifolds, Studies in Advanced Mathematics, Vol. 23, American Mathematical Society, Providence, RI, 2001, 151–182. [5] J. M. Maillard, Star exponential functions for any ordering of the elements of the inhomogeneous symplectic Lie algebra, to appear. [6] P. J. Olver, Non-associative local Lie groups, J. Lie Theory, 6 (1996), 23–59. [7] H. Omori, One must break symmetry in order to keep associativity, Banach Center Publ., 55 (2002), 1–11. [8] H. Omori, Beyond Point Set Topology, informal preprint for the Alanfest, Erwin Schrödinger Institute, Vienna, 2003. [9] H. Omori, Y. Maeda, N. Miyazaki, and A. Yoshioka, Strange phenomena related to ordering problems in quantizations, J. Lie Theory, 13-2 (2003), 481–510.

From momentum maps and dual pairs to symplectic and Poisson groupoids Charles-Michel Marle Institut de Mathématiques Université Pierre et Marie Curie 4, place Jussieu 75252 Paris Cedex 05 France [email protected] It is a great pleasure to submit a contribution for this volume in honour of Alan Weinstein. He is one of the four or five persons whose works have had the greatest influence on my own scientific interests, and I am glad to have this opportunity to express to him my admiration and my thanks.

Introduction In this survey, we will try to indicate some important ideas, due in large part to Alan Weinstein, which led from the study of momentum maps and dual pairs to the current interest in symplectic and Poisson groupoids. We hope that it will be useful for readers new to the subject; therefore, we begin by recalling the definitions and properties which will be used in what follows. More details can be found in [4, 26, 47]. 1. A Poisson manifold [27,E48] is a smooth manifold P equipped with a bivector field (i.e., a smooth section of 2 T P ) $ which satisfies [$, $] = 0, the bracket on the left-hand side being the Schouten bracket [44, 40]. The bivector field $ will be called the Poisson structure on P . It allows us to define a composition law on the space C ∞ (P , R) of smooth functions on P , called the Poisson bracket and denoted by (f, g) → {f, g}, by setting, for all f and g ∈ C ∞ (P , R) and x ∈ P , {f, g}(x) = $ df (x), dg(x) . That composition law is skew-symmetric and satisfies the Jacobi identity and therefore turns C ∞ (P , R) into a Lie algebra. 2. Let (P , $) be a Poisson manifold. We denote by $ : T ∗ P → T P the vector bundle map defined by

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C.-M. Marle

I J η, $ (ζ ) = $(ζ, η), where ζ and η are two elements in the same fibre of T ∗ P . Let f : P → R be a smooth function on P . The vector field Xf = $ (df ) is called the Hamiltonian vector field associated to f . If g : P → R is another smooth function on P , the Poisson bracket {f, g} can be written I J I J {f, g} = dg, $ (df ) = − df, $ (dg) . 3. Every symplectic manifold (M, ω) has a Poisson structure, associated to its symplectic structure, for which the vector bundle map $ : T ∗ M → M is the inverse of the vector bundle isomorphism v → −i(v)ω. We will always consider that a symplectic manifold is equipped with that Poisson structure, unless otherwise specified. 4. Let (P1 , $1 ) and (P2 , $2 ) be two Poisson manifolds. A smooth map ϕ : P1 → P2 is called a Poisson map if for every pair (f, g) of smooth functions on P2 , {ϕ ∗ f, ϕ ∗ g}1 = ϕ ∗ {f, g}2 . 5. The product P1 × P2 of two Poisson manifolds (P1 , $1 ) and (P2 , $2 ) has a natural Poisson structure: it is the unique Poisson structure for which the bracket of functions of the form (x1 , x2 ) → f1 (x1 )f2 (x2 ) and (x1 , x2 ) → g1 (x1 )g2 (x2 ), where f1 and g1 ∈ C ∞ (P1 , R), f2 and g2 ∈ C ∞ (P2 , R), is (x1 , x2 ) → {f1 , g1 }1 (x1 ){f2 , g2 }2 (x2 ). The same property holds for the product of any finite number of Poisson manifolds. 6. Let (V , ω) be a symplectic vector space, which means a real, finite-dimensional vector space V with a skew-symmetric nondegenrate bilinear form ω. Let W be a vector subspace of V . The symplectic orthogonal of W is K orth W = v ∈ V ; ω(v, w) = 0 for all w ∈ W }. It is a vector subspace of V , which satisfies dim W + dim(orth W ) = dim V ,

orth(orth W ) = W.

The vector subspace W is said to be isotropic if W ⊂ orth W , coisotropic if orth W ⊂ W , and Lagrangian if W = orth W . In any symplectic vector space, there are many Lagrangian subspaces; therefore, the dimension of a symplectic vector space is always even; if dim V = 2n, the dimension of an isotropic (resp., coisotropic, resp., Lagrangian) vector subspace is ≤ n (resp., ≥ n, resp., = n). 7. A submanifold N of a Poisson manifold (P , $) is said to be coisotropic if the bracket of two smooth functions, defined on an open subset of P and which vanish on N, vanishes on N too. A submanifold N of a symplectic manifold (M, ω) is coisotropic if and only if for each point x ∈ N , the vector subspace Tx N of the symplectic vector space Tx M, ω(x) is coisotropic. Therefore, the dimension of a coisotropic submanifold in a 2n-dimensional symplectic manifold is ≥ n; when it is equal to n, the submanifold N is said to be Lagrangian.

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8. A dual pair [48, 4] is a pair (ϕ1 : M → P1 , ϕ2 : M → P2 ) of smooth Poisson maps, defined on the same symplectic manifold (M, ω), with values in the Poisson manifolds (P1 , $1 ) and (P2 , $2 ), such that for each x ∈ M, the two equivalent equalities hold: ker(Tx ϕ1 ) = orth ker(Tx ϕ2 ) , ker(Tx ϕ2 ) = orth ker(Tx ϕ1 ) . That property implies that for all f1 ∈ C ∞ (P1 , R) and f2 ∈ C ∞ (P2 , R), {ϕ1∗ f1 , ϕ2∗ f2 } = 0. A dual pair (ϕ1 , ϕ2 ) is specially interesting when ϕ1 and ϕ2 are surjective submersions. 9. Let ϕ : M → P be a surjective submersion of a symplectic manifold (M, ω) onto a manifold P . The manifold P has a Poisson structure $ for which ϕ is a Poisson map if and only if orth(ker T ϕ) is integrable [23]. When that condition is satisfied, this Poisson structure on P is unique. If in addition there exist a smooth manifold P2 and a smooth map ϕ2 : M → P2 such that ker T ϕ2 = orth(ker T ϕ), the manifold P2 has a unique Poisson structure $2 for which ϕ2 is a Poisson map, and (ϕ, ϕ2 ) is a dual pair. 10. A symplectic realization [48] of a Poisson manifold (P , $) is a Poisson map ϕ : M → P , defined on a symplectic manifold (M, ω), with values in P . A symplectic realization ϕ : M → P is specially interesting when ϕ is a surjective submersion; such a symplectic realization is said to be surjective submersive. For example, in a dual pair (ϕ1 : M → P1 , ϕ2 : M → P2 ), ϕ1 and ϕ2 are symplectic realizations of the Poisson manifolds (P1 , $1 ) and (P2 , $2 ), respectively.

1 A typical example: action of a Lie group on its cotangent bundle Let G be a Lie group, πG : T ∗ G → G its cotangent bundle. For each g and h ∈ G, we write Lg (h) = gh, Rg (h) = hg. =g and R =g the canonical lifts to T ∗ G of Lg and Rg , respectively. We We denote by L recall that, for g and h ∈ G, ξ ∈ Th∗ G, X ∈ Tgh G and Y ∈ Thg G, we have I

J =g (ξ ), X = ξ, T Lg −1 X, L

I

J =g (ξ ), Y = ξ, T Rg −1 Y . R

=g ξ , and R = : T ∗ G × G → T ∗ G, = : G × T ∗ G → T ∗ G, (g, ξ ) → L The maps L =g ξ , are actions of the Lie group G on its cotangent bundle T ∗ G, on the (ξ, g) → R left and on the right, respectively. Theorem 1.1. These two actions are Hamiltonian and have as momentum maps, respectively, the maps JL : T ∗ G → G∗ ,

=π (ξ )−1 ξ JL (ξ ) = R G

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and

JR : T ∗ G → G ∗ ,

=π (ξ )−1 ξ, JR (ξ ) = L G

where G∗ is the dual of the Lie algebra G of G. We have identified G with Te G and G∗ with Te∗ G. We have denoted by πG : T ∗ G → G the cotangent bundle projection. Moreover, • • •

= the level sets of JL are the orbits of the action R, = the level sets of JR are the orbits of the action L, for each ξ ∈ T ∗ G, each one of the tangent spaces at ξ to the orbits of that point = and L = is the symplectic orthogonal of the other one. under the actions R

The dual G∗ of the Lie algebra G has two (opposite) natural Poisson structures, called the plus and the minus KKS-Poisson structures (the letters KKS stand for Kirillov [19], Kostant [21], and Souriau [45]). The brackets of two smooth functions f and g ∈ C ∞ (G∗ , R) are given by the formulae I

J I

J {f, g}+ (η) = η, df (η), dg(η) and {f, g}− (η) = − η, df (η), dg(η) . Then we have the following. Theorem 1.2. The map JL : T ∗ G → G∗ (resp., the map JR : T ∗ G → G∗ ) is a Poisson map when T ∗ G is equipped with the Poisson structure associated to its canonical symplectic structure and G∗ with the minus KKS-Poisson structure (resp, with the plus KKS-Poisson structure). The pair of maps (JL , JR ) in the above theorem is a very simple example of a dual pair; both JL and JR are surjective submersions. The cotangent space T ∗ G, equipped with its canonical structure, is a symplectic realization of each symplectic of the Poisson manifolds G∗ , {, }+ and G∗ , {, }− .

2 Hamiltonian action of a Lie group on a symplectic manifold The example dealt with in the preceding section is very symmetrical: the roles of the = and R = could be exchanged by means of the group anti-automorphism two actions L g → g −1 of the Lie group G. In this section, we will see that a similar situation (although less symmetrical) holds for a Hamiltonian action of a Lie group on a symplectic manifold. Definitions 2.1. Let : G × M → M be an action (for example, on the left) of a Lie group G on a symplectic manifold (M, ω). That action is said to be symplectic if, for any g ∈ G, ∗g ω = ω. It is said to be Hamiltonian if it is symplectic and if, in addition, there exists a smooth map J : M → G∗ such that, for each X ∈ G, vector field XM is I the fundamental J Hamiltonian, with the function J, X : x → J (x), X as Hamiltonian. The map J is called the momentum map of .


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2.2 Comments Let us indicate briefly some important properties of Hamiltonian actions. The fundamental vector fields Under the assumptions of the above definitions, we recall that the fundamental vector field XM associated to an element X ∈ G (the Lie algebra of G) is the vector field on M defined by d XM (x) = exp(tX), x t=0 , dt where x ∈ M. The formula i(XM )ω(x) = −dJ, X(x) expresses that XM is the Hamiltonian vector field associated to the function J, X. The momentum map equivariance When M is connected, there exists a smooth map θ : G → G∗ such that, for all g ∈ G and x ∈ M, J (g, x) = Ad ∗g J (x) + θ (g), where Ad ∗ : G × G∗ → G∗ is the coadjoint action, defined by I ∗ J I J Ad g (ξ ), X = ξ, Ad g −1 (X) , ξ ∈ G∗ , X ∈ G. The map θ satisfies, for all g and h ∈ G,

θ (gh) = Ad ∗g θ(h) + θ (g),

and is called a symplectic cocycle of G [45]. As a consequence, the map aθ : G × G ∗ → G ∗ ,

aθ (g, ξ ) = Ad ∗g (ξ ) + θ (g),

is an action on the left of G on G∗ , called the affine action associated to θ. The momentum map J : M → G∗ is equivariant when G acts on M by the action and on G∗ by the affine action aθ . The modified KKS-Poisson structures Moreover, the momentum map J is a Poisson map when M is equipped with the Poisson structure associated to its symplectic structure, and G∗ with the modified KKS-Poisson structure [45]: I

J {f, g}θ− (ξ ) = − ξ, df (ξ ), dg(ξ ) + ' df (ξ ), dg(ξ ) , where ' : G × G → R is the map defined by

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I J '(X, Y ) = Te θ (X), Y . When considered as a linear map from G to its dual G∗ , the map ' is a G∗ -valued 1cocycle of the Lie algebra G, which corresponds to the 1-cocycle θ of the Lie group G. Considered as a real-valued skew-symmetric bilinear map on G×G, ' is a real-valued 2-cocycle of the Lie algebra G. Symplectic orthogonality For M, each one of the vector subspaces of the symplectic vector space each x ∈ Tx M, ω(x) , • •

the tangent space at x to the orbit (G, x), the kernel of Tx J ,

is the symplectic orthogonal of the other one. 2.3 Remarks and questions Several features of dual pairs and symplectic realizations exist in a Hamiltonian action of a Lie group G on a symplectic manifold (M, ω): the momentum map J : M → G∗ is a symplectic realization of G∗ equipped with the modified KKS-Poisson structure; the symplectic orthogonality, for all x ∈ M, of ker Tx J and Tx (G, x), looks very much like the property of a dual pair; more precisely, if we assume that the set M/G of orbits of has a smooth manifold structure for which the canonical projection π : M → M/G is a submersion, there is on M/G a unique Poisson structure for which π is a Poisson map, and (J, π) is a dual pair. However, the momentum map J may not be a submersion (it is a submersion if and only if the action is locally free), and the set M/G may not have a smooth manifold structure for which π is a submersion. In order to make the Hamiltonian action of a Lie group more like the simple example of Section 1, we are led to the following questions: 1. Does there exist an “action’’ (in a generalized sense) on the manifold M whose orbits are the level sets of the momentum map J ? 2. In the theory of momentum maps, can we replace the dual of a Lie algebra by a more general Poisson manifold? 3. Does any Poisson manifold have a symplectic realization? The notion of symplectic groupoid, introduced in the next section, will allow us to answer some of these questions.

3 Lie groupoids and symplectic groupoids We recall below the definition of a groupoid. The reader will find examples and more information about groupoids in [4, 6, 33, 43, 52].


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Definition 3.1. A groupoid is a set equipped with the structure defined by the following data: • •

a subset 0 of , called the set of units of the groupoid; two maps α : → 0 and β : → 0 , called, respectively, the target map and the source map; they satisfy α|0 = β|0 = id 0 ;

•

a composition law m : 2 → , called the product, defined on the subset 2 of × , K L 2 = (x, y) ∈ × ; β(x) = α(y) , which is associative, in the sense that whenever one side of the equality m x, m(y, z) = m m(x, y), z

•

is defined, the other side is defined too, and the equality holds; moreover, the composition law m is such that for each x ∈ , m α(x), x = m x, β(x) = x; a map ι : → , called the inverse, such that, for every x ∈ , x, ι(x) ∈ 2 and ι(x), x ∈ 2 , and m x, ι(x) = α(x), m ι(x), x = β(x).

3.2 Properties and comments The above definitions have the following consequences. Involutivity of the inverse The inverse map ι is involutive. We have indeed, for any x ∈ , i 2 (x) = m i 2 (x), β i 2 (x) = m i 2 (x), β(x) = m i 2 (x), m i(x), x = m m i 2 (x), i(x) , x = m α(x), x = x. Unicity of the inverse Let x and y ∈ be such that m(x, y) = α(x)

and

m(y, x) = β(x).

Then we have y = m y, β(y) = m y, α(x) = m y, m x, ι(x) = m m(y, x), ι(x) = m β(x), ι(x) = m α ι(x) , ι(x) = ι(x). Therefore, for any x ∈ , the unique y ∈ such that m(y, x) = β(x) and m(x, y) = α(x) is ι(x).

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Notations A groupoid with set of units 0 and target and source maps α and β will be denoted α

by ⇒ 0 . β

When there is no risk of error, for x and y ∈ , we will write x.y, or even simply xy for m(x, y), and x −1 for ι(x). α

Definitions 3.3. A topological groupoid is a groupoid ⇒ 0 for which is a (maybe β

non-Hausdorff ) topological space, 0 a Hausdorff topological subspace of , α and β surjective continuous maps, m : 2 → a continuous map and ι : → an homeomorphism. α

A Lie groupoid is a groupoid ⇒ 0 for which is a smooth (maybe nonβ

Hausdorff ) manifold, 0 a smooth Hausdorff submanifold of , α and β smooth surjective submersions (which implies that 2 is a smooth submanifold of × ), m : 2 → a smooth map and ι : → a smooth diffeomorphism. 3.4 Properties and examples of Lie groupoids α

1. Let ⇒ 0 be a Lie groupoid. Since α and β are submersions, for any x ∈ , β α −1 α(x) and β −1 β(x) are submanifolds of , both of dimension dim −dim 0 , called the α-fibre and the β-fibre through x, respectively. The inverse map ι, restricted to the α-fibre through x (resp., the β-fibre through x) is a diffeomorphism of that fibre onto the β-fibre through ι(x) (resp., the α-fibre through ι(x)). The dimension of the submanifold 2 of composable pairs in × is 2 dim − dim 0 . 2. A Lie group is a Lie groupoid whose set of units has only one element e. 3. A vector bundle π : E → M is a Lie groupoid, with the base M as a set of units; the source and target maps both coincide with the projection π , the product and the inverse maps are the addition (x, y) → x + y and the opposite map x → −x in the fibres. α

4. Let ⇒ 0 be a Lie groupoid. Its tangent bundle T is a Lie groupoid, with T 0 β

as a set of units, T α : T → T 0 , and T β : T → T 0 as target and source maps. Let us denote by 2 the set of composable pairs in × , by m : 2 → the composition law and by ι : → the inverse. Then the set of composable pairs in T × T is simply T 2 , the composition law on T is T m : T 2 → T and the inverse is T ι : T → T . When the groupoid is a Lie group G, the Lie groupoid T G is a Lie group too. We will see below that the cotangent bundle of a Lie groupoid is a Lie groupoid, and more precisely a symplectic groupoid. Let us now introduce the important notion of symplectic groupoid, first considered by A. Weinstein [6], M. Karasev [18] and S. Zakrzewski [58].


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α

Definition 3.5. A symplectic groupoid is a Lie groupoid ⇒ 0 with a symplectic β

form ω on such that the graph of the composition law m K L (x, y, z) ∈ × × ; (x, y) ∈ 2 and z = m(x, y) is a Lagrangian submanifold of × × with the product symplectic form, the first two factors being endowed with the symplectic form ω, and the third factor being with the symplectic form −ω. The next theorem states important properties of symplectic groupoids. α

Theorem 3.6. Let ⇒ 0 be a symplectic groupoid, with the symplectic 2-form ω. β

We have the following properties: 1. For any point c ∈ , each one of the two vector subspaces of the symplectic vector space Tc , ω(c) , and Tc α −1 α(c) Tc β −1 β(c) is the symplectic orthogonal of the other one. 2 The submanifold of units 0 is a Lagrangian submanifold of the symplectic manifold (, ω). 3. The inverse map ι : → is an antisymplectomorphism of (, ω) (it satisfies ι∗ ω = −ω). Proof. For each x ∈ , we denote by Px = β −1 β(x) and Qx = α −1 α(x) the β-fibre and the α-fibre through x, respectively. Let dim = 2n. We have seen that dim 2 = 2 dim − dim 0 . Since the graph of the product is a Lagrangian submanifold of × × , its dimension is half that of × × , so 2(2 dim − dim 0 ) = 3 dim ; therefore, dim 0 = (1/2) dim = n. Since α and β are smooth submersions, for each point x ∈ , Px and Qx are smooth n-dimensional submanifolds of . 1. Let (a, b) ∈ 2 and c = m(a, b). The maps La : y → m(a, y) and Rb : x → m(x, b) are diffeomorphisms which map, respectively, Qb onto Qc and Pa onto Pc . Therefore, if u ∈ Ta Pa and v ∈ Tb Qb , w1 and w2 ∈ Tc , the vectors (u, 0, w1 ) and (0, v, w2 ) ∈ T(a,b,c) ( × × ) are tangent to the graph of the product m if and only if w1 = T Rb (u) and w2 = T La (v). By writing that the graph of m is Lagrangian in × × , we obtain ω(u, 0) + ω(0, v) − ω T Rb (u), T La (v) = 0, so, for all u ∈ Ta Pa and v ∈ Tb Qb ,

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ω(T Rb (u), T La (v) = 0. Since T Rb (u) can be any vector in Tc Pc and T La (v) any vector in Tc Qc , we have shown that orth(Tc Pc ) ⊃ Tc Qc . But since these two subspaces are of dimension n, orth(Tc Pc ) = Tc Qc , and orth(Tc Qc ) = Tc Pc . 2. Let p ∈ 0 . We have m(p, p) = p; therefore, for u1 and u2 ∈ Tp 0 , (u1 , u1 , u1 ) and (u2 , u2 , u2 ) are tangent to the graph of m. Since that graph is Lagrangian in × × , we have 0 = ω(u1 , u2 ) + ω(u1 , u2 ) − ω(u1 , u2 ) = ω(u1 , u2 ). This shows that 0 is an isotropic submanifold of . But since dim 0 = n, 0 is Lagrangian. 3. Let x ∈ , u1 and u2 ∈ Tx , v1 = T ι(u1 ), v2 = T ι(u2 ). Let t → s1 (t) and t →s2 (t) be smooth curves in such that s (0) = s (0) = x, ds1 (t)/dt |t=0 = u1 1 2 and ds2 (t)/dt |t=0 = u2 . For i = 1 or 2, we have m si (t), ι ◦ si (t) = α ◦ si (x). Therefore, if we set w1 = Tα(u1 ) and w2 = T α(u2 ), the vectors (u1 , v1 , w1 ) and (u2 , v2 , w2 ) are tangent at x, ι(x), α(x) to the graph of m. Since that graph is Lagrangian in × × , we have ω(u1 , u2 ) + ω T ι(u1 ), T ι(u2 ) − ω(w1 , w2 ) = 0. But since w1 and w2 are tangent at α(x) to the Lagrangian submanifold 0 , ω(w1 , w2 ) = 0. It follows that ι : → is an antisymplectomorphism.

α

Corollary 3.7. Let ⇒ 0 be a symplectic groupoid, with symplectic 2-form ω. There β

exists on 0 a unique Poisson structure $ for which α : → 0 is a Poisson map, and β : → 0 an anti-Poisson map (i.e., β is a Poisson map when 0 is equipped with the Poisson structure −$). The pair α : (, ω) → (0 , $), β : (, ω) → (0 , −$) is a dual pair, and (, ω) is a symplectic realization of both (0 , $) and (0 , −$). Proof. According to the previous theorem, the symplectic orthogonal of ker(T α) is ker(T β). By Property 9 of the Introduction, there exists on 0 a unique Poisson structure $ such that α is a Poisson map from (, ω) to (0 , $). For the same reason there exists on 0 another unique Poisson structure $ such that β is a Poisson map from (, ω) to (0 , $ ). But β = α ◦ ι, and the previous theorem shows that ι is an antisymplectomorphism. Therefore, $ = −$.

3.8 Cotangent bundle of a Lie groupoid α

Let ⇒ 0 be a Lie groupoid. We have seen above that its tangent bundle T has a β

Lie groupoid structure, determined by that of . Similarly (but much less obviously)


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the cotangent bundle T ∗ has a Lie groupoid structure determined by that of . The set of units is the conormal bundle to the submanifold 0 of , denoted by N∗ 0 . We recall that N∗ 0 is the vector subbundle of T∗0 (the restriction to 0 of the cotangent bundle T ∗ ) whose fibre Np∗ 0 at a point p ∈ 0 is K L Np∗ 0 = η ∈ Tp∗ ; η, v = 0 for all v ∈ Tp 0 . To define the target and source maps of the Lie algebroid T ∗ , we introduce the notion of bisection through a point x ∈ [6, 1, 4]. A bisection through x is a submanifold A of , with x ∈ A, transverse both to the α-fibres and to the β-fibres, such that the maps α and β, when restricted to A, are diffeomorphisms of A onto open subsets α(A) and β(A) of 0 , respectively. For any point x ∈ M, there exist bisections through x. A bisection A allows us to define two smooth diffeomorphisms between open subsets of , denoted by LA and RA and called the left and right translations by A, respectively. They are defined by LA : α −1 β(A) → α −1 α(A) , LA (y) = m β|−1 A ◦ α(y), y , and RA : β −1 α(A) → β −1 β(A) ,

RA (y) = m y, α|−1 A ◦ β(y) .

The definitions of the target and source maps for T ∗ rest on the following properties. Let x be a point in and let A be a bisection through x. The two vector subspaces, Tα(x) 0 and ker Tα(x) β, are complementary in Tα(x). Forany v ∈ Tα(x) , v −T β(v) is in ker Tα(x) β. Moreover, RA maps the fibre β −1 α(x) onto the fibre β −1 β(x) , and its restriction to that fibre does not depend on the choice of A; its depends only on x. Therefore, T RA v − T β(v) is in ker Tx β and does not depend on the choice of A. We can define the map = α by setting, for any ξ ∈ Tx∗ and any v ∈ Tα(x) , I J I J = α (ξ ), v = ξ, T RA v − T β(v) . = by setting, for any ξ ∈ Tx∗ and any w ∈ Tβ(x) , Similarly, we define β J I J I =(ξ ), w = ξ, T LA w − T α(w) . β = are unambiguously defined, smooth and take their values in the We see that = α and β ∗ submanifold N 0 of T ∗ . They satisfy π ◦ = α = α ◦ π ,

= = β ◦ π , π ◦ β

where π : T ∗ → is the cotangent bundle projection. Let us now define the composition law m = on T ∗ . Let ξ ∈ Tx∗ and η ∈ Ty∗ =(ξ ) = = be such that β α (η). That implies β(x) = α(y). Let A be a bisection through ∗ and a unique x and B a bisection through y. There exist a unique ξhα ∈ Tα(x) 0 ∗ ηhβ ∈ Tβ(y) 0 such that ∗ = ∗ ξ = (L−1 A ) β (ξ ) + αx ξhα ,

η = (RB−1 )∗ = α (ξ ) + βy∗ ηhβ .

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Then m =(ξ, η) is given by ∗ ∗ ∗ = m =(ξ, η) = αxy ξhα + βxy ηhβ + (RB−1 )∗ (L−1 A ) β (x) . =(ξ ) by = We observe that in the last term of the above expression we can replace β α (η), −1 ∗ −1 ∗ ∗ (R −1 )∗ , since these two expressions are equal, and that (RB ) (LA ) = (L−1 ) A B since RB and LA commute. Finally, the inverse= ι in T ∗ is ι∗ . = α

With its canonical symplectic form, T ∗ ⇒ N∗ 0 is a symplectic groupoid. = β

When the Lie groupoid is a Lie group G, the Lie groupoid T ∗ G is not a Lie group, contrary to what happens for T G. Its set of units can be identified with G∗ , = = JR . and we recover the typical example of Section 1, with = α = JL and β

4 Lie algebroids Let us now introduce the notion of a Lie algebroid, related to that of a Lie groupoid in the same way as the notion of a Lie algebra is related to that of a Lie group. That notion is due to J. Pradines [41]. Definition 4.1. A Lie algebroid over a smooth manifold M is a smooth vector bundle π : A → M with base M, equipped with • •

a composition law (s1 , s2 ) → {s1 , s2 } on the space ∞ (π ) of smooth sections of π, called the bracket, for which that space is a Lie algebra, a vector bundle map ρ : A → T M, over the identity map of M, called the anchor map, such that, for all s1 and s2 ∈ ∞ (π) and all f ∈ C ∞ (M, R), {s1 , f s2 } = f {s1 , s2 } + (ρ ◦ s1 ).f s2 .

4.2 Examples 1. A finite-dimensional Lie algebra is a Lie algebroid (with a base reduced to a point). 2. A tangent bundle τM : T M → M to a smooth manifold M is a Lie algebroid, with the usual bracket of vector fields on M as composition law, and the identity map as anchor map. More generally, any integrable vector subbundle F of a tangent bundle τM : T M → M is a Lie algebroid, still with the bracket of vector fields on M with values in F as composition law and the canonical injection of F into T M as anchor map. 3. Let X : M → T M be a smooth vector field on a smooth manifold M. By setting, for any pair (f, g) of smooth functions on M, [f, g] = f (X.g) − g(X.f ),


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we define on C ∞ (M, R) a composition law (which is a special case of a Jacobi bracket) which turns that space into a Lie algebra. We may identify the space C ∞ (M, R) of smooth functions on M with the space of smooth sections of the trivial vector bundle p1 : M × R → M, where p1 is the projection on the first factor; in that identification, a smooth function f ∈ C ∞ (M, R) is identified with the section sf : M → M × R, sf (x) = x, f (x) . The Jacobi bracket of functions defined above becomes a bracket (sf , sg ) → {sf , sg } = s[f,g] on the space of smooth sections of the trivial bundle p1 : M × R → M. It is easy to see that with the anchor map ρ : M × R → T M,

ρ(x, k) = kX(x),

that bundle becomes a Lie algebroid over M. 4. Let (P , $) be a Poisson manifold. Its cotangent bundle πP : T ∗ P → P has a Lie algebroid structure, with $ : T ∗ P → T P as anchor map. The composition law is the bracket of 1-forms, first obtained by Fuchssteiner [14], then independently by Magri and Morosi [36]. It will be denoted by (η, ζ ) → [η, ζ ] (in order to avoid any confusion with the Poisson bracket of functions). It is given by the formula, in which η and ζ are 1-forms and X a vector field on P , I J [η, ζ ], X = $ η, dζ, X + $ dη, X, ζ + L(X)$ (η, ζ ). We have denoted by L(X)$ the Lie derivative of the Poisson tensor $ with respect to the vector field X. Another equivalent formula for that composition law is [ζ, η] = L($ ζ )η − L($ η)ζ − d $(ζ, η) . The bracket of 1-forms is related to the Poisson bracket of functions by [df, dg] = d{f, g} for all f and g ∈ C ∞ (P , R). 4.3 Properties of Lie algebroids Let π : A → M be a Lie algebroid with anchor map ρ : A → T M. 1. It is easy to see that for any pair (s1 , s2 ) of smooth sections of π, ρ ◦ {s1 , s2 } = [ρ ◦ s1 , ρ ◦ s2 ], which means that the map s → ρ ◦ s is a Lie algebra homomorphism from the Lie algebra of smooth sections of π into the Lie algebra of smooth vector fields on M. 2. The composition law (s1 , s2 ) → {s1 , s2 } on the space of sections of π extends into a composition law on the space of sections of exterior powers of (A, π, M), which

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will be called the generalized Schouten bracket. Its properties are the same as those of the usual Schouten bracket [44, 40, 22]. When the Lie algebroid is a tangent bundle τM : T M → M, that composition law reduces to the usual Schouten bracket . When the Lie algebroid is the cotangent bundle πP : T ∗ P → P to a Poisson manifold (P , $), the generalized Schouten bracket is the bracket of forms of all degrees on the Poisson manifold P , introduced by J.-L. Koszul [22], which extends the bracket of 1 forms used in Example 4 of 4.2. 3. Let " : A∗ → M be the dual bundle of the Lie algebroid π : A → M. There exists on the space of sections of its exterior powers a graded endomorphism dρ , of E E degree 1 (this means that if η is a section of k A∗ , dρ (η) is a section of k+1 A∗ ). That endomorphism satisfies dρ ◦ dρ = 0, and its properties are essentially the same as those of the exterior derivative of differential forms. When the Lie algebroid is a tangent bundle τM : T M → M, dρ is the usual exterior derivative of differential forms. We can develop on the spaces of sections of the exterior powers of a Lie algebroid and of its dual bundle a differential calculus very similar to the usual differential calculus of vector and multivector fields and differential forms on a manifold [6, 4, 34, 37]. Operators such as the interior product, the exterior derivative and the Lie derivative can still be defined and have properties similar to those of the corresponding operators for vector and multivector fields and differential forms on a manifold. 4.4 The Lie algebroid of a Lie groupoid α

Let ⇒ 0 be a Lie groupoid. Let A() be the intersection of ker T α and T0 (the β

tangent bundle T restricted to the submanifold 0 ). We see that A() is the total space of a vector bundle π : A() → 0 , with base 0 , the canonical projection π being the map which associates a point u ∈ 0 to every vector in ker Tu α. We will define a composition law on the set of smooth sections of that bundle, and a vector bundle map ρ : A() → T 0 , for which π : A() → 0 is a Lie algebroid, callled α

the Lie algebroid of the Lie groupoid ⇒ 0 . β

We observe first that for any point u ∈ 0 and any point x ∈ β −1 (u), the map −1 y) Lx : y → Lx y = m(x, is defined on the α-fibre α (u), and maps that fibre −1 onto the α-fibre α α(x) . Therefore, Tu Lx maps the vector space Au = ker Tu α onto the vector space ker Tx α, tangent at x to the α-fibre α −1 α(x) . Any vector =(x) = w ∈ Au can therefore be extended into the vector field along β −1 (u), x → w Tu Lx (w). More generally, let w : U → A() be a smooth section of the vector bundle π : A() → 0 , defined on an open subset U of 0 . By using the above described construction for every point u ∈ U , we can extend the section w into a smooth vector field w =, defined on the open subset β −1 (U ) of , by setting, for all −1 u ∈ U and x ∈ β (u), w =(x) = Tu Lx w(u) .


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We have defined an injective map w → w = from the space of smooth local sections of π : A() → 0 , onto a subspace of the space of smooth vector fields defined on open subsets of . The image of that map is the space of smooth vector fields w =, defined = of of the form U = = β −1 (U ), where U is an open subset of 0 , on open subsets U which satisfy the two properties: (i) T α ◦ w = = 0, = such that β(x) = α(y), Ty Lx w (ii) for every x and y ∈ U =(y) = w =(xy). These vector fields are called left-invariant vector fields on . One can easily see that the space of left-invariant vector fields on is closed under the bracket operation. We can therefore define a composition law (w1 , w2 ) → {w1 , w2 } on the space of smooth sections of the bundle π : A() → 0 by defining {w1 , w2 } as the unique section such that {w w1 , w =2 ]. 1 , w2 } = [= Finally, we define the anchor map ρ as the map T β restricted to A(). One can easily check that with that composition law and that anchor map, the vector bundle π : A() → 0 is a Lie algebroid, called the Lie algebroid of the Lie groupoid α

⇒ 0 . β

We could exchange the roles of α and β and use right-invariant vector fields instead of left-invariant vector fields. The Lie algebroid obtained remains the same, up to an isomorphism. α

When the Lie groupoid ⇒ is a Lie group, its Lie algebroid is simply its Lie β

algebra. 4.5 The Lie algebroid of a symplectic groupoid α

Let ⇒ 0 be a symplectic groupoid, with symplectic form ω. As we have seen β

above, its Lie algebroid π : A → 0 is the vector bundle whose fibre, over each 0 point u ∈ 0 , is ker Tu α. We define a linear map ωu : ker Tu α → Tu∗ 0 by setting, for each w ∈ ker Tu α and v ∈ Tu 0 , I 0 J ωu (w), v = ωu (v, w). Since Tu 0 is Lagrangian and ker Tu α complementary to Tu 0 in the symplectic 0 vector space Tu , ω(u) , the map ωu is an isomorphism from ker Tu α onto Tu∗ 0 . By using that isomorphism for each u ∈ 0 , we obtain a vector bundle isomorphism of the Lie algebroid π : A → 0 onto the cotangent bundle π0 : T ∗ 0 → 0 . As seen in Corollary 3.7, the submanifold of units 0 has a unique Poisson structure $ for which α : → 0 is a Poisson map. Therefore, as seen in Example 4 of 4.2, the cotangent bundle π0 : T ∗ 0 → 0 to the Poisson manifold (0 , $) has a Lie

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algebroid structure, with the bracket of 1-forms as composition law. That structure is the same as the structure obtained as a direct image of the Lie algebroid structure of π : A() → 0 , by the above defined vector bundle isomorphism of π : A → 0 onto the cotangent bundle π0 : T ∗ 0 → 0 . The Lie algebroid of the symplectic α

groupoid ⇒ 0 can therefore be identified with the Lie algebroid π0 : T ∗ 0 → 0 , β

with its Lie algebroid structure of cotangent bundle to the Poisson manifold (0 , $). 4.6 The dual bundle of a Lie algebroid There exist some very close relationships between Lie algebroids and Poisson manifolds, discussed, for example, in [11]. We have already seen one such relationship: the cotangent bundle of a Poisson manifold has a Lie algebroid structure. We now describe another one. Let π : A → M be a Lie algebroid over a manifold M, with ρ : A → T M as anchor map. Let " : A∗ → M be the dual bundle of π : A → M. We observe that a smooth section s of π can be considered as a smooth function onI A∗ , whose J restriction to each fibre " −1 (x) (x ∈ M) is the linear function ζ → ζ, s(x) . By using that property, we see that the total space A∗ has a unique Poisson structure, whose bracket extends, for smooth functions, the bracket of sections of π . When the Lie algebroid is a finite-dimensional Lie algebra G, the Poisson structure on its dual space G∗ obtained by that means is the KKS-Poisson structure, already discussed in Section 1.

5 Integration of Lie algebroids and Poisson manifolds According to Lie’s third theorem, for any given finite-dimensional Lie algebra, there exists a Lie group whose Lie algebra is isomorphic to that Lie algebra. The same property is not true for Lie algebroids and Lie groupoids. The problem of finding necessary and sufficient conditions under which a given Lie algebroid is isomorphic to the Lie algebroid of a Lie groupoid remained open for more than 30 years. Partial results were obtained by J. Pradines [42], K. Mackenzie [33], P. Dazord [9], P. Dazord ans G. Hector [10]. A complete solution of that problem was obtained by M. Crainic and R. L. Fernandes [7]. Let us describe their very important work. 5.1 The Weinstein groupoid of a Lie algebroid Admissible paths in a Lie algebroid Let π : A → M be a Lie algebroid and ρ : A → T M its anchor map. Let a : I = [0, 1] → A be a smooth path in A. We will say that a is admissible if, for all t ∈ I , ρ ◦ a(t) =

d (π ◦ a)(t). dt


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We observe that when the Lie algebroid is the tangent bundle τM : T M → M, with the identity of T M as anchor map, a smooth path a : I → T M is admissible if and only if it is the canonical lift to T M of the smooth path τM ◦ a : I → M in M. For a general Lie algebroid, a smooth path a : I → A is admissible if and only if the map = a : T I = I × R → A,

= a (t, λ) = λa(t),

is a Lie algebroid homomorphism of the Lie algebroid p1 : I × R → I into the Lie algebroid π : A → M, over the map π ◦ a : I → M between the bases of these two Lie algebroids. Associated paths in a Lie groupoid and in its Lie algebroid Let us assume that π : A → M is the Lie algebroid of a Lie groupoid over M, α

⇒ M. Let γ : I = [0, 1] → be a smooth path in , starting from a unit β

x = γ (0) ∈ M ⊂ , and contained in the α-fibre α −1 (x), i.e., such that, for all t ∈ I , α ◦ γ (t) = x. dγ (t) is a vector tangent to the fibre α −1 (x), at the point γ (t). dt Applying to that vector a left translation by γ (t)−1 , we obtain a vector, dγ (t) aγ (t) = T Lγ (t)−1 ∈ ker Tβ◦γ (t) α. dt For each t ∈ I ,

But we have seen (4.4) that for each y ∈ M, the vector subspace ker Ty α of Ty is the α

fibre Ay over y of the Lie algebroid of the Lie groupoid ⇒ M. The map t → aγ (t) β

is therefore a smooth path in the Lie algebroid π : A → M. That path will be said to α

be associated to the path γ in the Lie groupoid ⇒ M. Since we have β

β ◦ Lγ (t)−1 = β, and since the anchor map of π : A → M is the restriction of T β, we see that the path aγ is admissible. Conversely, we see by integration that every smooth admissible path a in the Lie algebroid A is associated to a unique smooth path γ in the Lie groupoid , starting from the unit γ (0) = π ◦ a(0) ∈ M and contained in the α-fibre α −1 γ (0) . A Lie groupoid with connected and simply connected α-fibres We use the same assumptions as in the previous subsection. For smooth paths in starting from a unit in M and contained in an α-fibre, homotopy with fixed endpoints

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is an equivalence relation. The one-to-one correspondence γ → aγ , which associates, to each smooth path γ in starting from a unit and contained in an α-fibre, a smooth admissible path aγ in the Lie algebroid A, allows us to obtain an equivalence relation for smooth admissible paths in A. That equivalence relation will still be called homotopy. Let γ : I → and γ : I → be two smooth paths in such that, for all t ∈ I , γ (0) = α ◦ γ (t) = x ∈ M,

γ (0) = α ◦ γ (t) = y = β ◦ γ (1) ∈ M.

We can define a path γ .γ : I → by setting + γ (t) for 0 ≤ t ≤ 1/2, γ .γ (t) = γ (1).γ (2t − 1) for 1/2 ≤ t ≤ 1. That path starts from the unit x and is contained in the α-fibre α −1 (x). By replacing γ and γ by homotopic paths whose derivatives vanish on a neighbourhood of the endpoints 1 and 0, respectively, we may arrange things so that γ .γ is smooth (otherwise it is only piecewise smooth). By this means we obtain a composition law on the space of equivalence classes (for homotopy with fixed endpoints) of smooth paths in , starting from a unit and contained in an α-fibre. Crainic and Fernandes have shown [7] that this space, endowed with that composition law, is a Lie groupoid with connected and simply connected α fibres, and that the Lie algebroid of that Lie α

groupoid is π : A → M, the same as that of the Lie groupoid ⇒ M. Moreover, they β

show that that Lie groupoid is, up to an isomorphism, the unique Lie groupoid with connected and simply connected α-fibres whose Lie algebroid is π : A → M. That unicity property is the analogue of Lie’s firt theorem for Lie algebras and Lie groups. It was also proved by Moerdijk and Mrc˘ un [39] and by Mackenzie for transitive Lie algebroids [33]. Weinstein groupoid of a general Lie algebroid We no longer assume now that the Lie algebroid π : A → M is the Lie algebroid of a Lie groupoid. We cannot use any more paths in the groupoid , since may not exist, but we still can use admissible paths in the Lie algebroid A. As seen above, α

when π : A → M is the Lie algebroid of the Lie groupoid ⇒ M, homotopy with β

fixed endpoints for paths in starting from a unit and contained in an α-fibre induces an equivalence relation, still called homotopy, on the space of admissible paths in A. That equivalence relation can be expressed in terms involving the Lie algebroid π : A → M only, and still makes sense when that Lie algebroid is no longer the Lie algebroid of a Lie groupoid. That key observation allows us to consider the quotient of the space of smooth admissible paths in A by the homotopy equivalence relation. That quotient will be denoted by G(A). Crainic and Fernandes have shown that G(A) is endowed with a natural topological groupoid structure, and have called it the Weinstein


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groupoid of the Lie algebroid π : A → M (the idea of that construction being due to A. Weinstein). When that Lie algebroid is the Lie algebroid of a Lie groupoid, its Weinstein groupoid G(A) is a Lie groupoid, and is in fact the unique Lie groupoid with connected and simply connected α-fibres whose Lie algebroid is π : A → M. Conversely, Crainic and Fernandes have shown that when the topological groupoid G(A) is in fact a Lie groupoid, its Lie algebroid is isomorphic to π : A → M. The problem of finding necessary and sufficient conditions under which π : A → M is the Lie algebroid of a Lie groupoid amounts therefore to finding necessary and sufficient conditions under which the Weinstein groupoid G(A) is smooth, i.e., is a Lie groupoid. Crainic and Fernandes have solved that problem by introducing monodromy groups. 5.2 Monodromy groups Let π : A → M be a Lie algebroid, ρ : A → T M its anchor map and G(A) its Weinstein groupoid. For each x ∈ M, let Ax = π −1 (x), ρx = ρ|Ax and gx = ker ρx . Let u and v be two elements in gx , σu and σv two smooth sections of π : A → M such that σu (x) = u, σv (x) = v. The Leibniz rule shows that {σu , σv }(x) depends only on u and v, not on the sections σu and σv . This allows us to define the bracket [u, v] by setting [u, v] = {σu , σv }(x). With that bracket, gx is a Lie algebra. Let Nx (A) be the set of elements u in the center Z(gx ) of the Lie algebra gx such that the constant path t → u, t ∈ I = [0, 1], is equivalent (for the homotopy equivalence relation on the space of admissible smooth paths in A defined above) to the trivial path t → 0x , where 0x is the origin of the fibre Ax . Crainic and Fernandes have shown that Nx is a group, with the usual addition as composition law, which is at most countable, called the monodromy group at x. Let us take a Riemannian metric on the vector bundle π : A → M, and let d be the associated distance in the fibres of A. We set + d 0x , Nx (A) − {0x } if Nx (A) − {0x } = ∅, r(x) = +∞ if Nx (A) − {0x } = ∅. We see that r(x) > 0 if and only if the monodromy group Nx (A) is discrete. We may now state the main theorem. Theorem 5.3 (Crainic and Fernandes [7]). The Weinstein groupoid G(A) of the Lie algebroid π : A → M is a Lie groupoid if and only if the following two conditions are satisfied: (i) for all x ∈ M, the monodromy group Nx (A) is discrete, or in other words r(x) > 0; (ii) for all x ∈ M, we have lim inf r(y) > 0. y→x

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When these conditions are satisfied, the Lie algebroid π : A → M is said to be integrable. The reader will find in [7] several examples of Lie algebroids for which the monodromy groups are fully determined. There are Lie algebroids which are locally integrable (it means that any point in the base space of the Lie algebroid has an open neighbourhood such that when restricted to that neighbourhood, the Lie algebroid is integrable), but not globally integrable; in other words, integrability of Lie algebroids is not a local property. There are also Lie algebroids which are not locally integrable. 5.4 Applications and comments Integration of a Lie algebroid by a local Lie groupoid One may think of a local Lie groupoid as the structure defined on a smooth manifold by the following data: a smooth submanifold 0 ⊂ , smooth maps α, β, a composition law m and an inverse map ι, with the same properties as those of the corresponding maps of a Lie groupoid, but with the restriction that these maps are defined, and have these properties, only for elements in close enough to the space 0 of units. The Lie algebroid of a local Lie groupoid can be defined in the same way as that of a true Lie groupoid. J. Pradines [42] has shown that every Lie algebroid is the Lie algebroid of a local Lie groupoid. K. Mackenzie and P. Xu [35] have shown that when that Lie algebroid is the cotangent bundle to a Poisson manifold, the corresponding local Lie groupoid is a local symplectic groupoid. Crainic and Fernandes [7, 8] have shown that these results are now easy consequences of their general Theorem 5.3. Some integrable Lie algebroids By using Theorem 5.3, Crainic and Fernandes have proved the integrability of several types of Lie algebroids. Let us indicate some of their results A Lie algebroid with zero anchor map (i.e., a sheaf of Lie algebras) is always integrable, and the corresponding Lie groupoid is a sheaf of Lie groups (that result was already found by Douady and Lazard [12]). A regular Lie algebroid (i.e., a Lie algebroid whose anchor map is of constant rank) is locally integrable (but may be not globally integrable). A Lie algebroid whose anchor map is injective, or more generally injective on a dense open set, is integrable. 5.5 Symplectic realizations of a Poisson manifold The existence of local symplectic realizations of regular Poisson manifolds (i.e., with a Poisson structure of constant rank) was proved by Sophus Lie as early as 1890. The problem of finding a local symplectic realization of a Poisson manifold near a nonregular point is much more difficult. It was solved by Alan Weinstein in [48],


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where it is shown that if (P , $) is a Poisson manifold of dimension n and a ∈ P a point where the rank of $ is 2k, there exists a symplectic realization ϕ : M → U of an open neighbourhood U of a by a symplectic manifold M of dimension 2(n − k). Moreover, that realization is universal, in the sense that if ϕ : M → U is another symplectic realization of U , then dim M ≥ dim M and there exist (maybe after restriction of U and M ) a surjective Poisson submersion χ : M → M, whose fibres are symplectic submanifolds of M , such that ϕ = ϕ ◦ χ . By patching together symplectic realizations of open subsets of a Poisson manifold, A. Weinstein proved [49, 6] that any Poisson manifold has a global, surjective submersive symplectic realization. The same result was obtained independently by M. Karasev [18]. Another proof of that result was given by C. Albert and P. Dazord [1]. Weinstein and Karasev observed that such a realization automatically admits a local symplectic groupoid structure (this means a structure with a composition law, an inverse, source and target maps which look like those of a neighbourhood of the submanifold of units in a symplectic groupoid), the Poisson manifold being identified with the submanifold of units and the realization map either with the source or with the target map. The Lie algebroid of the (local) Lie groupoid obtained in that way can be identified with the cotangent bundle to the initially given Poisson manifold. The problem of finding a symplectic realization of a Poisson manifold (P , $) appears therefore as closely linked to the problem of finding a Lie groupoid whose Lie algebroid is the cotangent bundle T ∗ P , with the Lie algebroid structure described in Example 4 of 4.2. Integrable Poisson manifolds APoisson manifold (P , $) is said to be integrable if there exists a symplectic groupoid α

⇒ P , with P as submanifolds of units, the Poisson structure $ being that for which β

α is a Poisson map and β an anti-Poisson map. By using Theorem 5.3, Crainic and Fernandes have reinterpreted all known results about integrability of Poisson manifolds [8]. They have shown that a Poisson manifold (P , $) is integrable if and only if its cotangent bundle T ∗ P , with the Lie algebroid structure described in Example 4 of 4.2, is an integrable Lie algebroid. The symplectic groupoid which integrates (P , $) can be obtained as a symplectic quotient, as shown by Cattaneo and Felder [5]. They have shown that a Poisson manifold admits a complete realization if and only if it is integrable. 5.6 Examples Let us indicate the symplectic groupoids which can be associated to some examples of Poisson manifolds. 1. Let G∗ be the dual of a finite-dimensional Lie algebra G, with its KKS-Poisson structure. Let G be a Lie group with Lie algebra G. We can take as a symplectic groupoid associated to G∗ , the cotangent bundle T ∗ G with its natural Lie algebroid

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structure (described in 3.8). By choosing G connected and simply connected, we obtain a Lie groupoid structure on T ∗ G with connected and simply connected α- and β-fibres. 2. Let (M, ω) be a connected symplectic manifold. We can take as a symplectic groupoid associated to M (considered as a Poisson manifold) the product manifold M ×M, with the symplectic form p1∗ ω −p2∗ ω. We define on K M ×M the pair L groupoid structure, for which the set of units is the diagonal = (x, x); x ∈ M , identified with M. The target and source maps are α(x, y) = (x, x),

β(x, y) = (y, y),

x and y ∈ M.

But there is a better choice for the symplectic groupoid associated to M: the fundamental groupoid of M, denoted by $(M). It is the set of homotopy classes (with fixed ends) of smooth paths ϕ : [0, 1] → M. The set of units is now the set of homotopy classes of constant paths, which can be identified with M. The target and source maps associate, to the homotopy class = ϕ of a smooth path ϕ : [0, 1] → M, the homotopy classes of the constant paths equal to ϕ(0) and to ϕ(1), respectively. We have natural projections p1 : $(M) → M and p2 : $(M) → M, defined by p1 (= ϕ ) = ϕ(0) ϕ ) = ϕ(1). We take as a symplectic form on $(M) p1∗ ω − p2∗ ω. The fundaand p2 (= mental groupoid $(M) has, over the pair groupoid M × M, the advantage of having connected and simply connected α- and β-fibres. In the next section we describe a third example: the symplectic groupoid associated to a Poisson–Lie group.

6 Double symplectic groupoid of a Poisson–Lie group The notion of a Poisson–Lie group is due to Drinfel’d [13]. Let us recall its definition and some properties. The reader will find more details in [32, 50]. Definition 6.1. A Poisson–Lie group is a Lie group G, equipped with a Poisson structure $ such that the product m : G × G → G,

(x, y) → m(x, y) = xy

is a Poisson map (when G×G is equipped with the natural product Poisson structure). 6.2 Properties and examples 1. Any Lie group can be considered as a Poisson–Lie group, with the zero Poisson structure. 2. The Poisson tensor $ of a Poisson–Lie group G vanishes at the unit element e of G. The linearized Poisson structure at that point is a skew-symmetric composition law on Te∗ G which satisfies the Jacobi identity. Therefore, the dual G∗ of the Lie algebra G of G, which can be identified with Te∗ G, has a Lie algebra structure, determined by


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the Poisson structure on G. Therefore, we have a pair of vector spaces (G, G∗ ), each of these spaces being the dual of the other, both equipped with a Lie algebra structure. The pair (G, G∗ ) is called a Lie bialgebra. 3. The connected and simply connected Lie group G∗ with Lie algebra G∗ is called the dual Lie group of the Poisson–Lie group G. It also has a structure of Poisson–Lie group $∗ . When the Lie group G itself is connected and simply connected, the roles of G and G∗ are the same, they can be exchanged (in other words, the dual Lie group of the Poisson–Lie group (G∗ , $∗ ) is the Poisson–Lie group (G, $)). 4. On the vector space D = G ⊕ G∗ , there is a natural Lie algebra structure, of which G and G∗ are Lie subalgebras, whose bracket is [X1 + α1 , X2 + α2 ] = [X1 , X2 ] − ad ∗α2 X1 + ad ∗α1 X2 + [α1 , α2 ] + ad ∗X1 α2 − ad ∗X2 α1 , where X1 and X2 ∈ G, α1 and α2 ∈ G∗ . With that structure, D is called the double Lie algebra of G. 5. The connected and simply connected Lie group D with Lie algebra D is called the double Lie group of the Poisson–Lie group G. When G is assumed to be connected and simply connected, there exist natural injective Lie group homomorphisms G → D and G∗ → D, which will be denoted by g → g and u → u, respectively (with g ∈ G, u ∈ G∗ , g and u ∈ D). 6.3 Lu and Weinstein’s construction Let (G, $) be a connected and simply connected Poisson–Lie group (the assumption of simple connexity is made for simplicity, and can easily be removed). J.-H. Lu and A. Weinstein [31] have obtained a very nice description of a symplectic groupoid whose set of units is (G, $). We describe now that construction, with the above defined notations. Let K L = (g, u, v, h) ∈ G × G∗ × G∗ × G; gu = vh . Two different structures of Lie groupoid exist on , the first one with G as a set of units and the second one with G∗ as a set of units. We will denote by α1 , β1 , m1 and ι1 the target map, the source map, the composition law and the inverse map for the first structure, and by α2 , β2 , m2 and ι2 the corresponding maps for the second structure. They are given by the following formulae: α1 : (g, u, v, h) → (g, e, e, g), β1 : (g, u, v, h) → (h, e, e, h), m1 : (g1 , u1 , v1 , h1 = g2 ), (g2 = h1 , u2 , v2 , h2 ) → (g1 , u1 u2 , v1 v2 , h2 ), ι1 : (g, u, v, h) → (h, u−1 , v −1 , g), α2 : (g, u, v, h) → (e, v, v, e), β2 : (g, u, v, h) → (e, u, u, e), m2 : (g1 , u1 = v2 , v1 , h1 ), (g2 , u2 , v2 = u1 , h2 ) → (g1 g2 , u2 , v1 , h1 h2 ),

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ι2 : (g, u, v, h) → (g −1 , v, u, h−1 ). Moreover, has a symplectic structure ω compatible with each of its two Lie groupoid structures; in other words, with that symplectic structure, it is a symplectic groupoid in two different ways, with either G or G∗ as a set of units. Therefore, (, ω) is a symplectic realization of each of the two Poisson–Lie groups (G, $) and (G∗ , $∗ ).

7 Lie groupoid actions on a smooth manifold We have seen that not every pair of elements in a Lie groupoid can be composed: a pair (x, y) can be composed if and only if the image β(x), by the source map β, of the left element x, is equal to the image α(y), by the target map α, of the right element y. Similarly, to extend to a Lie groupoid action the well-known notion of a Lie group action on a smooth manifold, we must observe that not every pair made of an element in the groupoid and an element in the smooth manifold will be composable. For that reason, we need an extra ingredient, a map from the smooth manifold into the set of units of the goupoid, as shown in the following definition. α

Definition 7.1. Let ⇒ 0 be a Lie groupoid, M a smooth manifold and µ : M → 0 β

a smooth map. Let K L ×µ M = (x, m) ∈ × M; β(x) = µ(m) . We assume that ×µ M is a smooth submanifold of ×M. (This is true, for example, α

when µ is a submersion.) An action on the left of the Lie groupoid ⇒ 0 on the β

manifold M with moment map µ is a smooth map : ×µ M → M which satisfies the following properties: (i) µ (x, m) = α(x) for all (x, m) ∈ ×µ M, (ii) x, (y, m) = (xy, m) for all x and y ∈ , m ∈ M such that (x, y) ∈ 2 and (y, m) ∈ ×µ M, (iii) µ(m), m = m for all m ∈ M. A similar definition holds for an action on the right of a Lie groupoid on a smooth manifold. 7.2 Properties and examples α

1. A Lie groupoid ⇒ 0 acts on itself on the left with moment map α, and on on β

the right with moment map β. α

2. A Lie groupoid ⇒ 0 acts on both sides on the submanifold of units 0 , with β

moment map id 0 . These left and right actions are, respectively,


x, u = β(x) → α(xu) = α(x)

and

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u = α(x), x → β(ux) = β(x).

3. Property (ii) of the above definition implies that the moment map µ of a left action α

of a Lie groupoid ⇒ 0 on a smooth manifold M satisfies, for all x ∈ and β

m ∈ M such that β(x) = µ(m), µ (x, m) = α xµ(m) = α(x). In other words, the moment map µ is equivariant with respect to the left actions of α

the Lie groupoid ⇒ 0 on M and the left action of that groupoid on its submanifold β

of units 0 . A similar property holds for right actions. The following definition generalizes the notion of a symplectic (or Poisson) action of a Lie group on a symplectic (or Poisson) manifold. α

Definition 7.3. Let ⇒ 0 be a symplectic groupoid with symplectic form ω, (M, $) β

a Poisson manifold and µ : M → 0 a smooth map. Let : ×µ M → M be a α

smooth action of the Lie groupoid ⇒ 0 on the manifold M, with moment map µ. β

That action is called a Poisson action if its graph K L (x, m, p) ∈ × M × M; (x, m) ∈ ×µ M, p = (x, m) is a coisotropic submanifold of the product Poisson manifold × M × M, where is equipped with the Poisson structure associated to its symplectic structure, M with the Poisson structure $ and where M means the manifold M equipped with the Poisson structure −$. K. Mikami and A. Weinstein [38] have developed a theory of reduction for Poisson actions of symplectic groupoids very similar to the classical reduction theory for symplectic actions. The following proposition indicates an important property of the moment map for Poisson actions. Proposition 7.4. Let : ×µ M → M be a Poisson action of the symplectic α

groupoid ⇒ 0 on the Poisson manifold (M, $). The manifold of units 0 will be β

equipped with the unique Poisson structure for which the target map α : → 0 is a Poisson map. Then the moment map µ : M → 0 of that action is a Poisson map. Proof. Let s be a point in 0 , θ1 and θ2 ∈ Ts∗ 0 and n ∈ µ−1 (s). Let x ∈ , m ∈ M be such that β(x) = µ(m) and that (x, m) = n. Let ξ1 and ξ2 ∈ Tx∗ , η1 and η2 ∈ Tm∗ M and ζ1 and ζ2 ∈ Tn∗ M be such that (ξ1 , η1 , ζ1 ) and (ξ2 , η2 , ζ2 ) belong to the annihilator of the tangent space at (x, m, n)

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to the graph of . Since that graph is a coisotropic submanifold of × M × M, we have $ (ξ1 , ξ2 ) + $(η1 , η2 ) − $(ζ1 , ζ2 ) = 0. But by using the fact that µ ◦ = α ◦ p1 , where p1 : ×µ M → is the projection on the first factor, we see that (αx∗ θ1 , 0, −µ∗n θ1 ) and (αx∗ θ2 , 0, −µ∗n θ2 ) belong to the annihilator of the tangent space at (x, m, n) to the graph of . Therefore, $ (αx∗ θ1 , αx∗ θ2 ) − $(µ∗n θ1 , µ∗n θ2 ) = 0. But since α : → 0 is a Poisson map, $0 (θ1 , θ2 ) = $ (αx∗ θ1 , αx∗ θ2 ) = $(µ∗n θ1 , µ∗n θ2 ). That equality, which holds for all s ∈ 0 , θ1 and θ2 ∈ Ts∗ 0 and x ∈ µ−1 (s), proves that µ is a Poisson map. A shorter proof could be obtained by using the coisotropic calculus presented by A. Weinstein in [51], which extends to Poisson manifolds the calculus of symplectic relations initiated by W. M. Tulczyjew [46].

Conversely, P. Dazord [9] and P. Xu [55] have proved the following theorem. α

Theorem 7.5. Let ⇒ 0 be a local symplectic groupoid and (M, $) be a Poisson β

manifold. Every Poisson map µ : M → 0 is the momentum map for a unique α

α

β

β

local Poisson action of ⇒ 0 on (M, $). If ⇒ 0 is global (as a groupoid ), αconnected and α-simply connected, that action is global if and only if µ is a complete Poisson map. Let us explain some terms used in the above statement. The symplectic groupoid α

⇒ 0 is said to be α-connected and α-simply connected if the α-fibres are connected β

and simply connected. The moment map µ is said to be a complete Poisson map if for every smooth function f ∈ C ∞ (0 , R) whose Hamiltonian vector field on 0 is complete, the Hamiltonian vector field on M associated to the function µ∗ f = f ◦ µ is complete. 7.6 Example Let : G × M → M be a Hamiltonian action (on the left) of a Lie group G on a Poisson manifold (M, $), with an Ad ∗ -equivariant momentum map J : M → G∗ . α

Let T ∗ G ⇒ G∗ be the cotangent space of G, equipped with its canonical symplectic β

groupoid structure (3.8). Let K L T ∗ G ×J M = (ξ, m) ∈ T ∗ G × M; β(ξ ) = J (m) .


519

= : T ∗ G ×J M → M of that symplectic groupoid on the Poisson We define an action manifold (M, $), with moment map J , by setting, for all (ξ, m) ∈ T ∗ G ×J M, =(ξ, m) = πG (ξ ), m , where πG : T ∗ M → M is the canonical projection. That action is a Poisson action in the sense of Definition 7.3. This example shows that Hamiltonian actions of Lie groups, with Ad ∗ -equivariant momentum maps, appear as special cases of Poisson actions of symplectic groupoids. By a modification of the symplectic structure on T ∗ G, that result can be extended to Hamiltonian actions whose momentum map is not Ad ∗ -equivariant, but rather equivariant with respect to an affine action of G on G∗ . 7.7 Poisson actions of Poisson–Lie groups Let (G, $G ) be a Poisson–Lie group and (P , $P ) a Poisson manifold. An action on the left : G × P → P of the Lie group G on the manifold P is called a Poisson action if its graph K L (g, m, p) ∈ G × M × M; p = (g, m) is a coisotropic submanifold of the product Poisson manifold G × M × M, where M is the manifold M equipped with the Poisson structure −$. J.-H. Lu [30] has defined the notion of a momentum map for such an action. It is a map J : P → G∗ , with values in the dual Poisson–Lie group G∗ , such that, for each X in the Lie algebra G of G, XP = $P (J ∗ X r ),

where X r is the right-invariant 1-form on G∗ whose value at the unit element is X ∈ G (the vector space G being identified with the dual of Te G∗ , itself identified with G∗ ). A momentum map in the sense of Lu is a Poisson map. Along lines similar to those followed in 7.6, a Poisson–Lie group action on a Poisson manifold, with a momentum map in the sense of Lu, can be lifted to a Poisson action of the symplectic groupoid of G∗ .

8 Poisson groupoids Poisson groupoids were introduced by A. Weinstein [51] as a generalization of both symplectic groupoids and Poisson–Lie groups. α

Definition 8.1. A Poisson groupoid is a Lie groupoid ⇒ 0 , with a Poisson structure β

$ on , such that the graph of the product K L (x, y, z) ∈ × × ; (x, y) ∈ 2 , z = xy is a coisotropic submanifold of the product Poisson manifold × × , where is the manifold with the Poisson structure −$.

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8.2 Properties and examples 1. A symplectic groupoid is a Poisson groupoid whose Poisson structure is nondegenerate (i.e., symplectic). 2. A Poisson–Lie group is a Poisson groupoid whose groupoid structure is that of a Lie group (i.e., whose submanifold of units is reduced to one point). 3. As for a symplectic groupoid, the submanifold of units 0 of a Poisson groupoid α

⇒ 0 has a unique Poisson structure for which the maps α and β are, respectively, β

a Poisson and a anti-Poisson map. 4. The Lie algebroid π : A() → 0 of a Poisson groupoid has an additional structure: its dual bundle " : A()∗ → 0 also has a Lie algebroid structure, compatible in a certain sense (indicated below) with that of π : A() → 0 (K. Mackenzie and P. Xu [34], Y. Kosmann-Schwarzbach [20], Z.-J. Liu and P. Xu [29]). The compatibility condition between the two Lie algebroid structures on the two vector bundles in duality π : A → M and " : A∗ → M can be written as follows: d∗ [X, Y ] = L(X)d∗ Y − L(Y )d∗ X, where X and Y are two sections of π, or, using the generalized Schouten bracket (Property 2 of 4.3) of sections of exterior powers of the Lie algebroid π : A → M, d∗ [X, Y ] = [d∗ X, Y ] + [X, d∗ Y ]. In these formulae d∗ is the generalized exterior derivative, which acts on the space of sections of exterior powers of the bundle π : A → M, considered as the dual bundle of the Lie algebroid " : A∗ → M, defined in Property 3 of 4.3. These conditions are equivalent to the similar conditions obtained by exchange of the roles of A and A∗ . α When the Poisson groupoid ⇒ 0 is a symplectic groupoid, we have seen (4.5) β

that its Lie algebroid is the cotangent bundle π0 : T ∗ 0 → 0 to the Poisson manifold 0 (equipped with the Poisson structure for which α is a Poisson map). The dual bundle is the tangent bundle τ0 : T 0 → 0 , with its natural Lie algebroid structure defined in Property 2 of 4.2. 5. Conversely, K. Mackenzie and P. Xu [35] have shown that if the Lie algebroid of a Lie groupoid is a Lie bialgebroid (that means, if there exists on the dual vector bundle of that Lie algebroid a compatible structure of Lie algebroid, in the above defined sense), that Lie groupoid has a Poisson structure for which it is a Poisson groupoid. More information about Poisson groupoids can be found in [57].

9 Other developments Poisson geometry, symplectic and Poisson groupoids and their generalizations, are currently very active fields of research, and several aspects could not be discussed here.


521

Let us quote the works of S. Bates and A. Weinstein [3] on geometric quantization, of J. Huebschmann [15] and P. Xu [56] on Poisson cohomology, of J.-C. Marrero and D. Iglesias [16, 17] on Lie groupoids associated to Jacobi structures [28], of M. Bangoura and Y. Kosmann-Schwarzbach [2, 20] on the dynamical Yang–Baxter equation and Gerstenhaber algebras, of P. Libermann [24, 25] on contact groupoids and Lie algebroids. We refer to the excellent review papers of Alan Weinstein [53, 54] for a much more extensive survey and other references. Acknowledgments The author thanks the referee, who suggested important improvements upon the first version of that paper, and Ann Kostant for her patient help.

References [1] C. Albert and P. Dazord, Théorie des groupoïdes symplectiques: Chapitre II: Groupoïdes symplectiques, Publ. Dépt. Math. Univ. Claude Bernard Lyon I (N.S.), (1990), 27–99. [2] M. Bangoura and Y. Kosmann-Schwarzbach, Équation de Yang-Baxter dynamique classique et algébroïde de Lie, C. R. Acad. Sci. Paris Sér. I Math., 327 (1998), 541–546. [3] S. Bates and A. Weinstein, Lectures on the Geometry of Quantization, Berkeley Mathematics Lecture Notes, Vol. 8, American Mathematical Society, Providence, RI, 1997. [4] A. Cannas da Silva and A. Weinstein, Geometric Models for Noncommutative Algebras, Berkeley Mathematics Lecture Notes, Vol. 10, American Mathematical Society, Providence, RI, 1999. [5] A. S. Cattaneo and G. Felder, Poisson sigma models and symplectic groupoids, in Quantization of Singular Symplectic Quotients, Progress in Mathematics, Vol. 198, Birkhäuser, Boston, 2001, 41–73. [6] A. Coste, P. Dazord, and A. Weinstein, Groupoïdes symplectiques, Publ. Dépt. Math. Univ. Claude Bernard Lyon I (N.S.), 2/A (1987), 1–64. [7] M. Crainic and R. L. Fernandes, Integrability of Lie brackets, Ann. Math., 157 (2003), 575–620. [8] M. Crainic and R. L. Fernandes, Integrability of Poisson brackets, J. Differential Geom., 66-1, 71–137. November 2001. [9] P. Dazord, Groupoïdes symplectiques et troisième théorème de Lie “non linéaire,’’ in C. Albert, ed., Géombetrie Symplectique et Mécanique: Colloque International, La Grande Motte, France, 23–28 Mai, 1988, Lecture Notes in Mathematics, Vol. 1416, Springer-Verlag, Berlin, New York, Heidelberg, 1990, 39–74. [10] P. Dazord and G. Hector, Intégration symplectique des variétés de Poisson totalement asphériques, in P. Dazord and A. Weinstein eds., Symplectic Geometry, Groupoids, and Integrable Systems, Mathematical Sciences Research Institute Publications, Vol. 20, SpringerVerlag, New York, 1991, 37–72. [11] P. Dazord and D. Sondaz, Variétés de Poisson, Algébroïdes de Lie, Publ. Dépt. Math. Univ. Claude Bernard Lyon I (N.S.), 1/B (1988), 1–68. [12] A. Douady and M. Lazard, Espaces fibrés en algèbres de Lie et en groupes, Invent. Math., 1 (1966), 133–151. [13] V. G. Drinfel’d, Hamiltonian structures on Lie groups, Lie bialgebras and the geometric meaning of the classical Yang-Baxter equation, Soviet Math. Dokl., 27 (1983), 68–71. [14] B. Fuchssteiner, The Lie algebra structure of degenerate Hamiltonian and bi-Hamiltonian systems, Progr. Theoret. Phys., 68 (1982), 1082–1104.

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[15] J. Huebschmann, Poisson cohomology and quantization, J. Reine Angew. Math., 408 (1990), 57–113. [16] D. Iglesias Ponte, Lie Groups and Groupoids and Jacobi Structures, Thesis memory, Department of Fundamental Mathematics, Section of Geometry and Topology, Universidad de la Laguna, Spain, 2003. [17] D. Iglesias and J. C. Marrero, Generalized Lie bialgebroids and Jacobi structures, J. Geom. Phys., 40 (2001), 176–199. [18] M. Karasev, Analogues of the objects of Lie group theory for nonlinear Poisson brackets, Math. USSR Izvest., 28 (1987), 497–527. [19] A. Kirillov, Local Lie algebras, Russian Math. Surveys, 31 (1976), 55–75. [20] Y. Kosmann-Schwarzbach, Exact Gerstenhaber algebras and Lie bialgebroids, Acta Appl. Math., 41 (1995), 153–165. [21] B. Kostant, Quantization and unitary representations, in Lectures in Modern Analysis and Applications III, Lecture Notes in Mathematics, Vol. 170, Springer-Verlag, Berlin, 1970, 87–207. [22] J.-L. Koszul, Crochet de Schouten-Nijenhuis et cohomologie, Astérisque, hors série (1985), 257–271. [23] P. Libermann, Problèmes d’équivalence et géométrie symplectique, Astérisque, 107–108 (1983) (IIIe rencontre de géométrie du Schnepfenried, 10–15 Mai 1982, Vol. I), 43–68. [24] P. Libermann, On symplectic and contact groupoids, in O. Kowalski and D. Krupka, eds., Differential Geometry and Its Applications: Proceedings of the 5th International Conference, Opava, August 24–28, 1992, Silesian University, Opava, Czech Republic, 1993, 29–45. [25] P. Libermann, Lie algebroids and mechanics, Arch. Math., 32 (1996), 1147–162. [26] P. Libermann and Ch.-M. Marle, Symplectic Geometry and Analytical Mechanics, Kluwer, Dordrecht, the Netherlands, 1987. [27] A. Lichnerowicz, Les variétés de Poisson et leurs algèbres de Lie associées, J. Differential Geom., 12 (1977), 253–300. [28] A. Lichnerowicz, Les variétés de Jacobi et leurs algèbres de Lie associées, J. Math. Pures Appl., 57 (1978), 453–488. [29] Z.-J. Liu and P. Xu, Exact Lie algebroids and Poisson groupoids, Geom. Functional Anal., 6-1 (1996), 138–145. [30] J.-H. Lu, Momentum mappings and reduction of Poisson actions, in P. Dazord and A. Weinstein, eds., Symplectic Geometry, Groupoids, and Integrable Systems, Mathematical Sciences Research Institute Publications, Vol. 20, Springer-Verlag, New York, 1991, 209– 226. [31] J.-H. Lu and A. Weinstein, Groupoïdes symplectiques doubles des groupes de LiePoisson, C. R. Acad. Sci. Paris Sér. I Math., 309 (1989), 951–954. [32] J.-H. Lu and A. Weinstein, Poisson Lie groups, Dressing transformations and Bruhat decomposition, J. Differential Geom., 31 (1990), 501–526. [33] K. C. H. Mackenzie, Lie Groupoids and Lie Algebroids in Differential Geometry, London Mathmatical Society Lecture Notes, Vol. 124, Cambridge University Press, Cambridge, UK, 1987. [34] K. C. H. Mackenzie and P. Xu, Lie bialgebroids and Poisson groupoids, Duke Math. J., 73 (1994), 415–452. [35] K. C. H. Mackenzie and P. Xu, Integration of Lie bialgebroids, Topology, 39 (2000), 445–467. [36] F. Magri and C. Morosi, A Geometrical Characterization of Integrable Hamiltonian Systems through the Theory of Poisson-Nijenhuis Manifolds, Quaderno S 19, University of Milan, Milan, 1984.


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[37] C.-M. Marle, Differential calculus on a Lie algebroid and Poisson manifolds, in The J. A. Pereira da Silva Birthday Schrift, Textos de Matemática 32, Departamento de Matematica, Universidade de Coimbra, Coimbra, Portugal, 2002, 83-149. [38] K. Mikami and A. Weinstein, Moments and reduction for symplectic groupoid actions, Publ. RIMS Kyoto Univ., 24 (1988), 121–140. [39] I. Moerdijk and J. Mr˘cun, On integrability of infinitesimal actions, Amer. J. Math., 124 (2002), 567–593. [40] A. Nijenhuis, Jacobi-type identities for bilinear differential concomitants of certain tensor fields, Indag. Math., 17 (1955), 390–403. [41] J. Pradines, Théorie de Lie pour les groupoïdes différentiables: Calcul différentiel dans la catégorie des groupoïdes infinitésimaux, C. R. Acad. Sci. Paris Sér. A, 264 (1967), 245–248. [42] J. Pradines, Troisième théorème de Lie pour les groupoïdes différentiables, C. R. Acad. Sci. Paris Sér. A, 267 (1968), 21–23. [43] J. Renault, A Groupoid Approach to C ∗ -Algebras, Lecture Notes in Mathematics, Vol. 793, Springer-Verlag, Berlin, New York, Heidelberg, 1980. [44] J. A. Schouten, On the differential operators of first order in tensor calculus, in Convengo di Geometria Differenziale, Cremonese, Roma, 1953, 1–7. [45] J.-M. Souriau, Structure des Systèmes Dynamiques, Dunod, Paris, 1970. [46] W. M. Tulczyjew, Geometric Formulation of Physical Theories, Bibliopolis, Napoli, 1989. [47] I. Vaisman, Lectures on the Geometry of Poisson Manifolds, Birkhäuser, Basel, Boston, Berlin, 1994. [48] A. Weinstein, The local structure of Poisson manifolds, J. Differential Geom., 18 (1983), 523–557. [49] A. Weinstein, Symplectic groupoids and Poisson manifolds, Bull. Amer. Math. Soc., 16 (1987), 101–103. [50] A. Weinstein, Some remarks on dressing transformations, J. Fac. Sci. Univ. Tokyo Sect. IA Math., 35 (1988), 163–167. [51] A. Weinstein, Coisotropic calculus and Poisson groupoids, J. Math. Soc. Japan, 40 (1988), 705–727. [52] A. Weinstein, Groupoids: Unifying internal and external symmetry: A tour through some examples, Not. Amer. Math. Soc., 43 (1996), 744–752. [53] A. Weinstein, Poisson geometry, Differential Geom. Appl., 9 (1998), 213–238. [54] A. Weinstein, The Geometry of Momentum, 2002, arXiv: math.SG/0208108 v1. [55] P. Xu, Morita equivalence of Poisson manifolds, Comm. Math. Phys., 142 (1991), 493– 509. [56] P. Xu, Poisson cohomology of regular Poisson manifolds, Ann. Inst. Fourier Grenoble, 42-4 (1992), 967–988. [57] P. Xu, On Poisson groupoids, Internat. J. Math., 6-1 (1995), 101–124. [58] S. Zakrzewski, Quantum and classical pseudogroups I, II, Comm. Math. Phys., 134 (1990), 347–370, 371–395.

Construction of spectral invariants of Hamiltonian paths on closed symplectic manifolds∗ Yong-Geun Oh Department of Mathematics University of Wisconsin Madison, WI 53706 USA and Korea Institute for Advanced Study 207-43 Cheongnyangni 2-dong Dongdaemun-gu, Seoul 130-722 Korea [email protected] Dedicated to Alan Weinstein in honor of his 60th birthday. Abstract. In this paper, we develop a mini-max theory of the action functional over the semiinfinite cycles via the chain level Floer homology theory and construct spectral invariants of Hamiltonian paths on arbitrary, especially on nonexact and nonrational, compact symplectic manifold (M, ω). To each given time dependent Hamiltonian function H and quantum cohomology class 0 = a ∈ QH ∗ (M), we associate an invariant ρ(H ; a) which varies continuously over H in the C 0 -topology. This is obtained as the mini-max value over the semiinfinite cycles whose homology class is “dual’’ to the given quantum cohomology class a on the covering 0 (M) of the contractible loop space 0 (M). We call them the Novikov Floer cycles. space We apply the spectral invariants to the study of Hamiltonian diffeomorphisms in sequels of this paper. We assume that (M, ω) is strongly semipositive here, to be removed in a sequel to this paper.

1 Introduction and main results The group Ham(M, ω) of (compactly supported) Hamiltonian diffeomorphisms of the symplectic manifold (M, ω) carries a remarkable invariant norm defined by φ = inf H H →φ

H =

1

(1.1) (max Ht − min Ht )dt

0 ∗ This research was partially supported by the NSF grant DMS-9971446, by NSF grant DMS-

9729992 at the Institute for Advanced Study, by a Vilas Associate Award at the University of Wisconsin, and by a grant of the Korean Young Scientist Prize.

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which was introduced by Hofer [Ho]. Here H → φ means that φ is the time-one map 1 of the Hamilton equation x˙ = X (x) of the Hamiltonian H : [0, 1] × M → R, φH H where the Hamiltonian vector field is defined by ω(XH , ·) = dH.

(1.2)

This norm can be easily defined on arbitrary symplectic manifolds although proving nondegeneracy is a nontrivial matter (See [Ho, Po1, LM] for its proof of increasing generality. See also [Ch] for a Floer-theoretic proof and [Oh3] for a simple proof of the nondegeneracy in tame symplectic manifolds). On the other hand Viterbo [V] defined another invariant norm on R2n . This was defined by considering the graph of the Hamiltonian diffeomorphism φ : R2n → R2n and compactifying the graph in the diagonal direction in R4n = R2n ×R2n into T ∗ S 2n . He then applied the critical point theory of generating functions of the Lagrangian submanifold, graph φ ⊂ T ∗ S 2n , which he developed on the cotangent bundle T ∗ N of the arbitrary compact manifold N . To each cohomology class a ∈ H ∗ (N ), Viterbo associated certain homologically essential critical values of generating functions of any Lagrangian submanifold L Hamiltonian isotopic to the zero section of T ∗ N and proved that they depend only on the Lagrangian submanifold but not on the generating functions, at least up to normalization. The present author [Oh1, Oh2] and Milinkovic´ [MO1, MO2, Mi] developed a Floer-theoretic approach to the construction of Viterbo’s invariants using the canonically defined action functional on the space of paths, utilizing the observation made by Weinstein [W] that the action functional is a generating function of the given Lagrangian submanifold defined on the path space. This approach is canonical including normalization and provides a direct link between Hofer’s geometry and Viterbo’s invariants in a transparent way. One of the key points in our construction in [Oh2] is the emphasis on the usage of the existing group structure on the space of Hamiltonians defined by t −1 (H, K) → H #K := H + K ◦ (φH ) (1.3) in relation to the pants product and the triangle inequality. However, we failed to fully exploit this structure and fell short of proving the triangle inequality at the time of writing [Oh1, Oh2]. This construction can be carried out for the Hamiltonian diffeomorphisms as long as the action functional is single valued, e.g., on weakly-exact symplectic manifolds. Schwartz [Sc] carried out this construction in the case of symplectically aspherical (M, ω), i.e., for (M, ω) with c1 |π2 (M) = ω|π2 (M) = 0. Among other things he proved the triangle inequality for the invariants constructed using the notion of Hamiltonian fibration and (flat) symplectic connection on it. It turns out that the proof of this triangle inequality [Sc] is closely related to the notion of the K-area of the Hamiltonian fibration [Po2] with connections [GLS, Po2], especially to the one with fixed monodromy studied by Entov [En1]. In this context, the choice of the triple (H, K; H #K) we made in [Oh2] can be interpreted as the one which makes infinity the K-area of the corresponding Hamiltonian fibration over the Riemann surface of genus zero with three punctures equipped with the given monodromy around the

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punctures. Entov [En1] develops a general framework of Hamiltonian connections with fixed boundary monodromy and relates the K-area with various quantities of the given monodromy which are of the Hofer length type. This framework turns out to be particularly useful for our construction of spectral invariants in this paper. On nonexact symplectic manifolds, the action functional is not single valued and the Floer homology theory has been developed as a circle-valued Morse theory or a 0 (M) of the space 0 (M) of contractible (free) Morse theory on a covering space loops on M in the literature related to Arnold’s conjecture which was initiated by Floer himself [Fl]. The Floer theory now involves quantum effects and uses the Novikov ring in an essential way [HoS]. The presence of quantum effects and denseness of the action spectrum in R (as in nonrational symplectic manifolds), had been the most serious obstacle that has plagued the study of the family of Hamiltonian diffeomorphisms, until the author [Oh4] developed a general framework of the mini-max theory over 0 (M) which we call the Novikov natural semiinfinite cycles on the covering space Floer cycles. In this paper, we will exploit the “finiteness’’ condition in the definitions of the Novikov ring and the Novikov Floer cycles in a crucial way for the proofs of various existence results of pseudoholomorphic curves that are needed in the proofs of the axioms of spectral invariants and nondegeneracy of the norm that we construct [Oh8]. Although the Novikov ring is essential in the definition of the Floer homology and the quantum cohomology in the literature, as far as we know it is the first time for the finiteness condition to be explicitly used beyond the purpose of giving the definition of the quantum cohomology and the Floer homology. A brief description of the setting of the Floer theory [HoS] is in order, partly to fix our convention: Let (γ , w) be a pair of γ ∈ 0 (M) and w a disc bounding γ . We say that (γ , w) is -equivalent to (γ , w ) iff ω([w #w]) = 0 and

c1 ([w #w]) = 0,

(1.4)

where w is the map with opposite orientation on the domain and w #w is the obvious glued sphere. Here stands for the group =

π2 (M) . ker(ω|π2 (M) ) ∩ ker(c1 |π2 (M) )

0 (M) the set of We denote by [γ , w] the -equivalence class of (γ , w) and by 0 (M) → 0 (M) be the canonical projection. We -equivalence classes. Let π : 0 (M) the -covering space of 0 (M). The action functional A0 : 0 (M) → R call is defined by A0 ([γ , w]) = −

w∗ ω.

(1.5)

Two -equivalent pairs (γ , w) and (γ , w ) have the same action and so the action is 0 (M). When a one-periodic Hamiltonian H : (R/Z) × M → R is well defined on (M) → R by given, we consider the functional AH : ∗ (1.6) AH ([γ , w]) = − w ω − H (t, γ (t))dt.

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Our convention is chosen to be consistent with the classical mechanics Lagrangian on the cotangent bundle with the symplectic form ω0 = −dθ, θ = pi dq i i

when (1.2) is adopted as the definition of Hamiltonian vector field. See the remark in the end of this introduction on other conventions in the symplectic geometry. The conventions in this paper coincide with our previous papers [Oh1, Oh2, Oh4] and Entov’s [En1, En2] but different from many other literature on the Floer homology in some ways. (There was a sign error in [Oh1, Oh2] when we compare the Floer complex and the Morse complex for a small Morse function, which was rectified in [Oh4]. In our convention, the positive gradient flow of f corresponds to the negative gradient flow of Af .) The mini-max theory of this action functional on the -covering space has been implicitly used in the proof of Arnold’s conjecture. Recently, the author has further developed this mini-max theory via the Floer homology and applied it to the study of Hofer’s geometry of Hamiltonian diffeomorphism groups [Oh4]. We also outlined construction of spectral invariants of Hamiltonian diffeomorphisms of the type [V, Oh2, Sc] on arbitrary nonexact symplectic manifolds for the classical cohomological classes. The main purpose of this paper is to further develop the chain level Floer theory introduced in [Oh4] and to carry out construction of spectral invariants for arbitrary quantum cohomology classes. The organization of the paper is now in order. In Section 2, we briefly review various facts related to the action functional and its action spectrum. Some of these may be known to the experts, but precise details for 0 (M) of general (M, ω) first appeared the action functional on the covering space in our paper [Oh5] especially concerning the normalization and the loop effect on the action spectrum: We define the action spectrum of H by 0 (M), dAH ([z, w]) = 0}, Spec(H ) := {AH ([z, w]) ∈ R | [z, w] ∈ 0 (M) → R. In [Oh5], we have shown that i.e., the set of critical values of AH : once we normalize the Hamiltonian H on compact M by Ht dµ = 0 M

with dµ the Liouville measure, Spec(H ) depends only on the equivalence class = [φ, H ] (see Section 2 for the definition) and so Spec(φ ) ⊂ R is a well-defined φ subset of R for each φ ∈ Ham(M, ω). Here π : Ham(M, ω) → Ham(M, ω) is the universal covering space of Ham(M, ω). This kind of normalization of the action spectrum is a crucial point for systematic study of the spectral invariants of the Viterbo type in general. Schwarz [Sc] previously proved that in the aspherical case

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where the action functional is single valued already on 0 (M), this normalization can be made on Ham(M, ω), not just on Ham(M, ω). In Section 3, we review the quantum cohomology and its Morse theory realization of the corresponding complex. We emphasize the role of the Novikov ring in relating the quantum cohomology and the Floer homology and the reversal of upward and downward Novikov rings in this relation. In Section 4, we review the standard operators in the Floer homology theory and explain the filtration naturally present in the Floer complex and how it changes under the Floer chain map. In Section 5, we give the definition of our spectral invariants for the Hamiltonian functions H , and prove finiteness of the mini-max values ρ(H ; a). In Section 6, we prove all the basic properties of the spectral invariants. We summarize these into the following theorem. We ∞ ([0, 1] × M) the set of normalized continuous functions on [0, 1] × M. denote by Cm ∞ ([0, 1] × M) and Noting that there is a one–one correspondence between the set Cm the set of Hamiltonian paths t λ = φH : t ∈ [0, 1] → φH ∈ Ham(M, ω),

one may equally consider ρ(H ; a) as an invariant attached to the Hamiltonian path φH . Theorem I. Let (M, ω) be arbitrary closed symplectic manifold. For any given quantum cohomology class 0 = a ∈ QH ∗ (M), we have a continuous function denoted by ∞ ρ = ρ(H ; a) : Cm ([0, 1] × M) × QH ∗ (M) → R ∞ ([0, 1] × M) be smooth such that they satisfy the following axioms: Let H, F ∈ Cm ∗ Hamiltonian functions and a = 0 ∈ QH (M). Then ρ satisfies the following axioms:

(1) Projective invariance: ρ(H ; λa) = ρ(H ; a) for any 0 = λ ∈ Q. (2) Normalization: For a = A∈ aA q −A , we have ρ(0; a) = v(a), where 0 is the zero function and v(a) := min{ω(−A) | aA = 0} = − max{ω(A) | aA = 0}

(1.7)

is the (upward ) valuation of a. (3) Symplectic invariance: ρ(η∗ H ; a) = ρ(H ; a) for any symplectic diffeomorphism η. (4) Triangle inequality: ρ(H #F ; a · b) ≤ ρ(H ; a) + ρ(F ; b). (5) C 0 -continuity: |ρ(H ; a) − ρ(F ; a)| ≤ H #F = H − F , where · is the ∞ ([0, 1] × M). In particular, the function ρ : H → Hofer’s pseudonorm on Cm a 0 ρ(H ; a) is C -continuous. We will call the set spec(H ) := {ρ(H ; a) | a ∈ QH ∗ (M)}

(1.8)

the essential spectrum of H . Most of the properties stated in this theorem are direct analogues to the ones in [Oh1, Oh2, Sc]. Except for the proof of finiteness of ρ(H ; a), proofs of all of the

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properties are refinements of the arguments used in [Oh2, Oh4, Sc]. In addition, the proof of the triangle inequality uses the concept of Hamiltonian fibration with fixed monodromy and the K-area [Po2, En1], which is an enhancement of the arguments used in [Oh2, Sc]. In the classical mini-max theory for the indefinite functionals [Ra, BnR], there was implicitly used the notion of “semiinfinite cycles’’ to carry out the mini-max procedure. There are two essential ingredients needed to prove existence of actual critical values out of the mini-max values: one is the finiteness of the mini-max value, or the linking property of the (semiinfinite) cycles associated to the class a and the other is to prove that the corresponding mini-max value is indeed a critical value of the action functional. When the global gradient flow of the action functional exists as in the classical critical point theory [BnR], this point is closely related to the well-known Palais–Smale condition and the deformation lemma which are essential ingredients needed to prove the criticality of the mini-max value. Partly because we do not have the global flow, we need to geometrize all these classical mini-max procedures. It turns out that the Floer homology theory in the chain level is the right framework for this purpose. In Section 7, we will restrict to the rational case and prove the following additional property of spectral invariants, the spectrality axiom. We will study the nonrational cases elsewhere for which we expect the same property holds, at least for the nondegenerate Hamiltonian functions, but its proof seems to be much more nontrivial. We now recall the definition of rational symplectic manifolds: Denote ω := {ω(A) | A ∈ π2 (M)} = ω() ⊂ R and Spec(H ) = ∪z∈Per(H ) Spec(H ; z). Recall that ω is either a discrete or a countable dense subset of R. Definition 1.1. A symplectic manifold (M, ω) is called rational if ω is discrete. Theorem II (spectrality axiom). Suppose that (M, ω) be rational. Then ρ satisfies the following additional properties: (1) For any smooth one-periodic Hamiltonian function H : S 1 × M → R, we have ρ(H ; a) ∈ Spec(H ) for each given quantum cohomology class 0 = a ∈ QH ∗ (M). (2) For two smooth functions H ∼ K, we have ρ(H ; a) = ρ(K; a)

(1.9)

for all a ∈ QH ∗ (M). In particular, ρ can be pushed down to the “universal covering space’’ Ham(M, ω) of Ham(M, ω) by putting ρ(φ ; a) to be the this common value for φ = [H ]. We call ) ⊂ Spec(φ ) defined by the subset spec(φ

Spectral invariants

531

) = {ρ(φ ; a) | a ∈ QH ∗ (M)} spec(φ . Then we have the following refined the (homologically) essential spectrum of φ version of Theorem II for the rational cases. Theorem III. Let (M, ω) be rational and define the map ρ : Ham(M, ω) × QH ∗ (M) → R ; a) := ρ(H ; a). Let φ , ψ ∈ Ham(M, by ρ(φ ω) and a = 0 ∈ QH ∗ (M). Then ρ satisfies the following axioms: ; a) ∈ Spec(φ ). (1) Spectrality: For each a ∈ QH ∗ (M), ρ(φ (2) Projective invariance: ρ( φ ; λa) = ρ(φ ; a) for any 0 = λ ∈ Q. (3) Normalization: For a = A∈ aA q −A , we have ρ(0; a) = v(a), where 0 is the identity in Ham(M, ω) and v(a) := min{ω(−A) | aA = 0} = − max{ω(A) | aA = 0}

(1.10)

is the (upward ) valuation of a. ; a) for any symplectic diffeomorη−1 ; a) = ρ(φ (4) Symplectic invariance: ρ(ηφ phism η. · ψ ; a · b) ≤ ρ(φ ; a) + ρ(ψ ; b). (5) Triangle inequality: ρ(φ ; a) − ρ(ψ ; a)| ≤ φ ◦ ψ −1 , where · is the Hofer’s (6) C 0 -continuity: |ρ(φ → ρ(φ ; a) is pseudonorm on Ham(M, ω). In particular, the function ρa : φ 0 C -continuous. act on Ham(M, (7) Monodromy shift: Let [h, h] ∈ π0 (G) ω)×QH ∗ (M) by the map , a) → (h · φ , (φ h∗ a), where h∗ a is the image of the (adjoint) Seidel’s action [Se] by [h, h] on the quantum cohomology QH ∗ (M). Then we have , a)) = ρ(φ ; a) + Iω ([h, ρ([h, h] · (φ h]).

(1.11)

It would be an interesting question to ask whether these axioms characterize the spectral invariants ρ. It is related to the question whether the graph of the sections → ρ(φ ; a); ρa : φ

Ham(M, ω) → Spec(M, ω)

can be split into other “branch’’ in a way that the other branch can also satisfy all the above axioms or not. Here the action spectrum bundle Spec(M, ω) is defined by A ) ⊂ Ham(M, Spec(M, ω) := Spec(φ ω) × R. ∈H φ am(M,ω)

We will investigate this question elsewhere.

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To get the main stream of ideas in this paper without getting bogged down with technicalities related with transversality question of various moduli spaces, we assume in this paper that (M, ω) is strongly semipositive in the sense of [Se, En1]: A closed symplectic manifold is called strongly semipositive if there is no spherical homology class A ∈ π2 (M) such that ω(A) > 0,

2 − n ≤ c1 (A) < 0.

Under this condition, the transversality problem concerning various moduli spaces of pseudoholomorphic curves is standard. We will not mention this generic transversality question at all in the main body of the paper unless it is absolutely necessary. In Section 8, we will briefly explain how this general framework can be incorporated in our proofs in the context of Kuranishi structure [FOn] all at once. In the appendix, we introduce the notion of continuous quantum cohomology and explain how to extend our definition of spectral invariants to the continuous quantum cohomology classes. This work originated from a part of our paper entitled “Mini-max theory, spectral invariants and geometry of the Hamiltonian diffeomorphism group’’ [Oh6] that has been circulated since July, 2002. We isolate and streamline the construction part of spectral invariants from [Oh6] in this paper with some minor corrections and addition of more details. In particular, we considerably simplify the definition of ρ(H ; a) from [Oh6] here. We leave the application part of [Oh6] to a separate paper [Oh8] in which we construct the homological norm of Hamiltonian diffeomorphism and apply them to the study of geometry of Hamiltonian diffeomorphisms on general compact symplectic manifolds. Another application of the spectral invariants to the study of length minimizing property of Hamiltonian paths is given by the author [Oh7, Oh8]. See also [En2, EnP] for other interesting applications of spectral invariants. In another sequel to this paper, we will provide a description of spectral invariants in terms of the Hamiltonian fibration. Convention (1) The Hamiltonian vector field Xf associated to a function f on (M, ω) is defined by df = ω(Xf , ·). (2) The addition F #K and the inverse K on the set of time periodic Hamiltonians C ∞ (M × S 1 ) are defined by F #G(x, t) = F (x, t) + G((φFt )−1 (x), t), t G(x, t) = −G(φG (x), t).

There is another set of conventions which are used in the literature (e.g., in [Po3]): (1) Xf is defined by ω(Xf , ·) = −df (2) The action functional has the form AH ([z, w]) = −

w∗ ω +

H (t, z(t))dt.

(1.12)

Spectral invariants

533

Because our Xf is the negative of Xf in this convention, the action functional is the one for the Hamiltonian −H in our convention. While our convention makes the positive Morse gradient flow correspond to the negative Cauchy–Riemann flow, the other convention keeps the same direction. The reason we keep our convention is that we would like to keep the definition of the action functional the same as the classical Hamilton functional pdq − H dt (1.13) on the phase space and to make the negative gradient flow of the action functional for the zero Hamiltonian become the pseudoholomorphic equation. It appears that the origin of the two different conventions is the choice of the convention as to how one defines the canonical symplectic form on the cotangent bundle T ∗ N or in the classical phase space: If we set the canonical Liouville form pi dq i θ= i

for the canonical coordinates q 1 , . . . , q n , p1 , . . . , pn of T ∗ N , we take the standard symplectic form to be ω0 = −dθ = dq i ∧ dpi , while the people using the other convention (see, e.g., [Po3]) take ω0 = dθ = dpi ∧ dq i . As a consequence, the action functional (1.12) in the other convention is the negative of the classical Hamilton functional (1.13). It seems that there is not a single convention that makes everybody happy and hence one has to live with some nuisance in this matter one way or the other.

2 The action functional and the action spectrum Let (M, ω) be any compact symplectic manifold and let 0 (M) be the set of con0 (M) be its the covering space mentioned before. We will always tractible loops and consider normalized functions f : M → R by f dµ = 0, (2.1) M

where dµ is the Liouville measure of (M, ω). When a periodic normalized Hamiltonian H : M × (R/Z) → R is given, we (M) → R by consider the action functional AH : AH ([γ , w]) = − w∗ ω − H (γ (t), t)dt. We denote by Per(H ) the set of periodic orbits of XH .

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Definition 2.1. We define the action spectrum of H , denoted as Spec(H ) ⊂ R, by 0 (M), z ∈ Per(H )}, Spec(H ) := {AH (z, w) ∈ R | [z, w] ∈ (M) → R. For each given z ∈ Per(H ), we i.e., the set of critical values of AH : denote Spec(H ; z) = {AH (z, w) ∈ R | (z, w) ∈ π −1 (z)}. Note that Spec(H ; z) is a principal homogeneous space modeled by the period group of (M, ω) ω := {ω(A) | A ∈ π2 (M)} = ω() ⊂ R and Spec(H ) = ∪z∈Per(H ) Spec(H ; z). The following was proved in [Oh4]. Lemma 2.2. For any closed symplectic manifold (M, ω) and for any smooth Hamiltonian H , Spec(H ) is a measure zero subset of R for any H . For given φ ∈ Ham(M, ω), we denote F → φ if φF1 = φ, and denote H(φ) = {F | F → φ}. We say that two Hamiltonians F and K are equivalent and denote F ∼ K if they are connected by one parameter family of Hamiltonians {F s }0≤s≤1 such that F s → φ for all s ∈ [0, 1]. We write [F ] for the equivalence class of F . Then the universal (étale) covering space Ham(M, ω) of Ham(M, ω) is realized by the set of such equivalence classes. Note that the group G := (Ham(M, ω), id) of based loops naturally acts on the loop space (M) by (h · γ )(t) = h(t)(γ (t)), where h ∈ (Ham(M, ω)) and γ ∈ (M). An interesting consequence of Arnold’s conjecture is that this action maps 0 (M) to itself (see, e.g., [Se, Lemma 2.2]). Seidel 0 (M). The set of lifts (h, [Se, Lemma 2.4] proves that this action can be lifted to h) forms a covering group G → G ⊂ G × Homeo( 0 (M)) G whose fiber is isomorphic to . Seidel relates the lifting (h, h) of h : S 1 → Ham(M, ω) to a section of the Hamiltonian bundle associated to the loop h (see [Se, Section 2]). When a Hamiltonian H generating the loop h is given, the assignment z → h · z provides a natural one–one correspondence

Spectral invariants

h : Per(F ) → Per(H #F ),

535

(2.2)

t )−1 . Let F, K be normalized Hamiltonians with where H #F = H + F ◦ (φH F, K → φ and let H be the Hamiltonian such that K = H #F , and ft , gt , and ht the corresponding Hamiltonian paths as above. In particular, the path h = {ht }0≤t≤1 defines a loop. We also denote the corresponding action of h on 0 (M) by h. Let h 0 (M)). Then a straightforward calculation shows (see be any lift of h to Homeo( [Oh5]) that h∗ (dAF ) = dAK (2.3)

0 (M). In particular, since 0 (M) is connected, we have as a one-form on h∗ (AF ) − AK = C(F, K, h),

(2.4)

where C = C(F, K, h) is a constant a priori depending on F, K, h. Theorem 2.3 ([Oh5, Theorem II]). Let h be the loop as above and h be a lift. Then the constant C(F, K, h) in (2.4) depends only on the homotopy class [h, h] ∈ π0 (G). In particular, if F ∼ K, we have AF ◦ h = AK and hence Spec F = Spec K ∈ Ham(M, as a subset of R. For any φ ω), we define ) := Spec F Spec(φ . for a (and so any) normalized Hamiltonian F with [φ, F ] = φ Definition 2.4 (action spectrum bundle). We define the action spectrum bundle of (M, ω) by A Spec(M, ω) = Specφ(M, ω) ⊂ Ham(M, ω) × R, ∈H φ am(M,ω)

where = [F ]} ⊂ R Specφ(M, ω) = {AF ([z, w]) | dAF ([z, w]) = 0, φ and denote by π : Spec(M, ω) → Ham(M, ω) the natural projection.

3 Quantum cohomology in the chain level We first recall the definition of the quantum cohomology ring QH ∗ (M). As a module, it is defined as QH ∗ (M) = H ∗ (M, Q) ⊗ ↑ω , ↑

where ω is the (upward) Novikov ring

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Y.-G. Oh

+ ↑ω

=

aA q

−A

| aA ∈ Q, # A | ai = 0,

A∈

−A

3 ω < λ < ∞ ∀λ ∈ R .

Due to the finiteness assumption on the Novikov ring, we have the natural (upward) valuation v : QH ∗ (M) → R defined by ⎛ ⎞ v⎝ aA q −A ⎠ = min{ω(−A) : aA = 0} (3.1) A∈ω

which for any a, b ∈ QH ∗ (M) satisfies that v(a + b) ≥ min{v(a), v(b)}. Definition 3.1. For each homogeneous element a = A∈ aA q −A ∈ QH k (M),

aA ∈ H ∗ (M, Q),

(3.2)

of degree k, we also call v(a) the level of a and the corresponding term in the sum the leading order term of a and denote by σ (a). Note that the leading order term σ (a) of a homogeneous element a is unique among the summands in the sum by the definition (1.4) of . The product on QH ∗ (M) is defined by the usual quantum cup product, which we denote by “·’’ and which preserves the grading, i.e., satisfies QH k (M) × QH (M) → QH k+ (M). Often the homological version of the quantum cohomology is also useful, sometimes called the quantum homology, which is defined by QH∗ (M) = H∗ (M) ⊗ ↓ω , ↓

where ω is the (downward) Novikov ring ⎧ ⎫ + 3 ⎨ ⎬ ↓ω = bj q Bj | bj ∈ Q, # Bj | bj = 0, ω > λ < ∞ ∀λ ∈ R . ⎩ ⎭ Bj Bj ∈

We define the corresponding (downward) valuation by ' * B v = max{ω(B) : aB = 0} aB q B∈

which for f, g ∈ QH∗ (M) satisfies that v(f + g) ≤ max{v(f ), v(g)}.

(3.3)

Spectral invariants

537

↓

We like to point out that the summand in ω is written as bB q B while the one in ↑ ω as aA q −A with the minus sign. This is because we want to clearly show which one we use. Obviously −v in (3.1) and v in (3.3) satisfy the axiom of non-Archimedean norm which induce a topology on QH ∗ (M) and QH∗ (M), respectively. In each case the finiteness assumption in the definition of the Novikov ring allows us to numerate the nonzero summands in each given Novikov chain (3.2) so that λ1 > λ2 > · · · > λj > · · · → −∞ with λj = ω(Bj ) or ω(Aj ). Since the downward Novikov ring appears mostly in this paper, we will just use ω ↓ or for ω , unless absolutely necessary to emphasize the direction of the Novikov ring. We define the level and the leading order term of b ∈ QH∗ (M) similarly as in Definition 3.1 by changing the role of upward and downward Novikov rings. We have a canonical isomorphism 0 : QH ∗ (M) → QH∗ (M); ai q −Ai → P D(ai )q Ai and its inverse : QH∗ (M) → QH ∗ (M);

bj q Bj →

P D(bj )q −Bj .

We denote by a 0 and b# the images under these maps. There exists the canonical nondegenerate pairing ·, · : QH ∗ (M) ⊗ QH∗ (M) → Q defined by

M

ai q −Ai ,

N (ai , bj )δAi Bj , bj q Bj =

(3.4)

where δAi Bj is the delta function and (ai , bj ) is the canonical pairing between H ∗ (M, Q) and H∗ (M, Q). Note that this sum is always finite by the finiteness condition in the definitions of QH ∗ (M) and QH∗ (M) and so is well defined. This is equivalent to the Frobenius pairing in the quantum cohomology ring. However, we would like to emphasize that the dual vector space (QH∗ (M))∗ of QH∗ (M) is not isomorphic to QH ∗ (M) even as a Q-vector space. Rather the above pairing induces an injection QH ∗ (M) → (QH∗ (M))∗ whose images lie in the set of continuous linear functionals on QH∗ (M) with respect to the topology induced by the valuation v. (3.3) on QH∗ (M). We refer to [Br] for a good introduction to non-Archimedean analytic geometry. In fact, the description of the standard quantum cohomology in the literature is not really a “cohomology’’ but a “homology’’ in that it never uses linear functionals in its definition. To keep our exposition consistent with the standard literature in the Gromov–Witten invariants and quantum cohomology, we prefer to call them the quantum cohomology rather

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than quantum homology as some authors did (e.g., [Se]) in the symplectic geometry community. In the appendix, we will introduce a genuinely cohomological version of quantum cohomology which we call continuous quantum cohomology using the continuous linear functionals on the quantum chain complex below with respect to the topology induced by the valuation v. Let (C∗ , ∂) be any chain complex on M whose homology is the singular homology H∗ (M). One may take for C∗ the usual singular chain complex or the Morse chain complex of a Morse function f : M → R, (C∗ (−f ), ∂−f ) for some sufficiently small > 0. However, since we need to take a nondegenerate pairing in the chain level, we should use a model which is finitely generated. We will always prefer to use the Morse homology complex because it is finitely generated and avoids some technical issue related to singular degeneration problem of the type studied in [FOh1, FOh2]. The negative sign in (C∗ (−f ), ∂−f ) is used to make the correspondence between the Morse homology and the Floer homology consistent with our conventions of the Hamiltonian vector field (1.2) and the action functional (1.6). In our conventions, solutions of the negative gradient of −f correspond to those for the negative gradient flow of the action functional Af . We denote by (C ∗ (−f ), δ−f ) the corresponding cochain complex, i.e., C k := Hom(Ck , Q),

∗ δ−f = ∂−f .

Now we extend the complex (C∗ (−f ), ∂−f ) to the quantum chain complex, denoted by (CQ∗ (−f ), ∂Q ) CQ∗ (−f ) := C∗ (−f ) ⊗ ω ,

∂Q := ∂−f ⊗ ω .

(3.5)

This coincides with the Floer complex (CF∗ (f ), ∂) as a chain complex if is sufficiently small. Similarly, we define the quantum cochain complex (CQ∗ (−f ), δ Q ) by changing the downward Novikov ring to the upward one. In other words, we define CQ∗ (−f ) := CM2n−∗ (−f ) ⊗ ↑ ,

δ Q := ∂f ⊗ ↑ω .

Again we would like to emphasize that CQ∗ (−f ) is not isomorphic to the dual space of CQ∗ (−f ) as a Q-vector space. We refer to the appendix for some further discussion on this issue. It is well known that the corresponding homology of this complex is independent of the choice f and isomorphic to the above quantum cohomology (respectively, the quantum homology) as a ring (see [PSS, LT2, Lu] for its proof). This isomorphism, however, plays no significant role in the current paper, except as a bookkeeping device for the family of invariants ρ(H ; a) that we associate to each quantum cohomology class a ∈ QH ∗ (M) later. (See Section 5.1 for more explanation about this point.) To emphasize the role of the Morse function in the level of complex, we denote the corresponding homology by H Q∗ (−f ) ∼ = QH ∗ (M).

Spectral invariants

539

With these definitions, we have the obvious nondegenerate pairing CQ∗ (−f ) ⊗ CQ∗ (−f ) → Q

(3.6)

in the chain level which induces the pairing (3.4) above in homology. We now choose a generic Morse function f . Then for any given homotopy H = {H s }s∈[0,1] with H 0 = f and H 1 = H , we denote by hH : CQ∗ (−f ) = CF∗−n (f ) → CF∗−n (H )

(3.7)

the standard Floer chain map from f to H via the homotopy H. This induces a homomorphism hH : H Q∗ (−f ) ∼ = H F∗−n (f ) → H F∗−n (H ).

(3.8)

Although (3.7) depends on the choice H, (3.8) is canonical, i.e., does not depend on the homotopy H. One confusing point in this isomorphism is the issue of grading. See the next section for a review of the construction of this chain map and the issue of grading of H F∗ (H ).

4 Filtered Floer homology For each given generic nondegenerate H : S 1 × M → R, we consider the free Q vector space over 0 (M) | z ∈ Per(H )}. Crit AH = {[z, w] ∈

(4.1)

To be able to define the Floer boundary operator correctly, we need to complete this vector space downward with respect to the real filtration provided by the action AH ([z, w]) of the element [z, w] of (4.1). More precisely, we have the following. Definition 4.1. We call the formal sum β= a[z,w] [z, w],

a[z,w] ∈ Q

(4.2)

[z,w]∈Crit AH

a Novikov chain if there are only finitely many nonzero terms in the expression (4.2) above any given level of the action. We denote by CF∗ (H ) the set of Novikov chains. We call those [z, w] with a[z,w] = 0 generators of the chain β and just denote as [z, w] ∈ β in that case. Note that CF∗ (H ) is a graded Q-vector space which is infinite dimensional in general, unless π2 (M) = 0. As in [Oh4], we introduce the following notion which is a crucial concept for the mini-max argument we carry out later.

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Y.-G. Oh

Definition 4.2. Let β be a Novikov chain in CF∗ (H ). We define the level of the cycle β and denote by λH (β) = max{AH ([z, w]) | a[z,w] = 0 in (4.2)} [z,w]

if β = 0, and we put λH (0) = −∞ as usual. We call the unique critical point [z, w] that realizes the maximum value λH (β) the peak of the cycle β, and denote it by pk(β). We briefly review construction of basic operators in the Floer homology theory [Fl]. Let J = {Jt }0≤t≤1 be a periodic family of compatible almost complex structure on (M, ω). For each given pair (J, H ), we define the boundary operator ∂ : CF∗ (H ) → CF∗ (H ) considering the perturbed Cauchy–Riemann equation + ∂u ∂u ∂τ + J ∂t − XH (u) = 0, limτ →−∞ u(τ ) = z− , limτ →∞ u(τ ) = z+ .

(4.3)

0 (M), defines nothing but the negative gradient flow This equation, when lifted to 0 (M) induced by the family of metrics on M of AH with respect to the L2 -metric on gJt = (·, ·)Jt := ω(·, Jt ·): This L2 -metric is defined by

1

ξ, ηJ := 0

(ξ, η)Jt dt.

We will also denote v2J0 = (v, v)J0 = ω(v, J0 v)

(4.4)

for v ∈ T M. For each given [z− , w− ] and [z+ , w+ ], we define the moduli space M(H, J ; [z− , w− ], [z+ , w+ ]) of solutions u of (4.3) with finite energy ' 2 * ∂u 2 ∂u 1 + dtdτ < ∞ EJ (u) = ∂τ ∂t − XH (u) 1 2 R×S

and satisfying

Jt

w − #u ∼ w+ .

∂ has degree −1 and satisfies ∂ ◦ ∂ = 0.

Jt

(4.5)

Spectral invariants

541

When we are given a family (j, H) with H = {H s }0≤s≤1 and j = {J s }0≤s≤1 , the chain homomorphism h(j,H) : CF∗ (H 0 ) → CF∗ (H 1 ) is defined by the nonautonomous equation + ∂u ρ1 (τ ) ∂u − X H ρ2 (τ ) (u) = 0, ∂τ + J ∂t limτ →−∞ u(τ ) = z− , limτ →∞ u(τ ) = z+

(4.6)

also with the condition (4.5). Here ρi , i = 1, 2 is the cutoff functions of the type ρ : R → [0, 1], + 0 for τ ≤ −R, ρ(τ ) = 1 for τ ≥ R, ρ (τ ) ≥ 0 for some R > 0. h(j,H) has degree 0 and satisfies ∂(J 1 ,H 1 ) ◦ h(j,H) = h(j,H) ◦ ∂(J 0 ,H 0 ) . Two such chain maps for different homotopies (j 1 , H1 ) and (j 2 , H2 ) connecting the same endpoints are also known to be chain homotopic [Fl]. Finally, when we are given a homotopy (j , H) of homotopies with j = {jκ }, H = {Hκ }, consideration of the parameterized version of (4.6) for 0 ≤ κ ≤ 1 defines the chain homotopy map HH : CF∗ (H 0 ) → CF∗ (H 1 ),

(4.7)

which has degree +1 and satisfies h(j1 ,H1 ) − h(j0 ,H0 ) = ∂(J 1 ,H 1 ) ◦ HH + HH ◦ ∂(J 0 ,H 0 ) .

(4.8)

By now, construction of these maps using these moduli spaces has been completed with rational coefficients (see [FOn, LT1, Ru]) using the techniques of virtual moduli cycles. We will suppress this advanced machinery from our presentation throughout the paper. The main stream of the proof is independent of this machinery except that it is implicitly needed to prove that various moduli spaces we use are nonempty. Therefore, we do not explicitly mention these technicalities in the main body of the paper until Section 8, unless it is absolutely necessary. In Section 8, we will provide justification of this in the general case all at once. The following upper estimate of the action change can be proved by the same argument as used in the proof of [Ch, Oh1, Oh4]. We would like to emphasize that in general there does not exist a lower estimate of this type. The upper estimate is just one manifestation of the “positivity’’ phenomenon in symplectic topology through the existence of pseudoholomorphic curves first discovered by Gromov [Gr]. On the other

542

Y.-G. Oh

hand, the existence of lower estimate is closely tied to some nontrivial homological property of (Floer) cycles, and best formulated in terms of Floer cycles instead of individual critical points [z, w] for the nondegenerate Hamiltonians. However, we would like to point out that the equations (4.3) and (4.6) or the numerical estimate of the action changes for solutions u with finite energy can be studied for any H or (H, j ) which are not necessarily nondegenerate or generic, although the Floer complex or the operators may not be defined for such choices. Proposition 4.3. Let H, F be any Hamiltonian not necessarily nondegenerate and j = {J s }s∈[0,1] be any given homotopy and let Hlin = {H s }0≤s≤1 be the linear homotopy H s = (1 − s)H + sF . Suppose that (4.6) has a solution satisfying (4.5). Then we have the identity AF ([z+ , w+ ]) − AH ([z− , w− ]) 2 ∞ ∂u = − − ρ (τ )(F (t, u(τ, t)) − H (t, u(τ, t)))dtdτ (4.9) ∂τ J ρ1 (τ ) −∞ 2 1 ∂u ≤ − + − min (Ft − Ht )dt (4.10) x∈M ∂τ J ρ1 (τ ) 0 1 ≤ − min (Ft − Ht )dt. (4.11) 0

x∈M

By considering the case F = H , we immediately have the following. Corollary 4.4. For a fixed H and for a given one parameter family j = {J s }s∈[0,1] , let u be as in Proposition 4.3. Then we have AH ([z+ , w+ ]) − AH ([z− , w− ]) = −

2 ∂u ∂τ ρ (τ ) ≤ 0. J 1

(4.12)

Remark 4.5. We would like to remark that similar calculation proves that there is also an uniform upper bound C(j, H) for the chain map over general homotopy (j, H) or for the chain homotopy maps (4.7). In this case, the identity (4.9) is replaced by AF ([z+ , w+ ]) − AH ([z− , w− ]) 2 ∞ ∂u ∂H s =− − ρ (τ ) (t, u(τ, t)) dtdτ ∂τ J ρ1 (τ ) ∂s s=ρ(τ ) −∞ 2 1 ∂u ∂H s ≤ − + − min dt x∈M ∂τ J ρ1 (τ ) ∂s s=ρ(τ ) 0 1 ∂Hts ≤ − min dt. (4.13) x∈M ∂s 0 This upper estimate is also crucial for the construction of these maps. This upper estimate depends on the choice of homotopy (j, H) and is related to the curvature estimates of the relevant Hamiltonian fibration (see [Po2, En1]).

Spectral invariants

543

Now we recall that CF∗ (H ) is also a -module: each A ∈ acts on Crit AH , and so on CF∗ (H ) by “gluing a sphere’’ A : [z, w] → [z, w#A]. Then ∂ is -linear and induces the standard Floer homology H F∗ (H ; ) with as its coefficients (see [HoS] for a detailed discussion on the Novikov ring and on the Floer complex as a -module). However, the action does not preserve the filtration we defined above. Whenever we talk about filtration, we will always presume that the relevant coefficient ring is Q. For a given nondegenerate H and an λ ∈ R \ Spec(H ), we define the relative chain group CFkλ (H ) := {β ∈ CFk (H ) | λH (β) < λ}. Corollary 4.4 implies that between the two chain complexes (CFk (H ), ∂(H,J ) ) and (CFk (H ), ∂(H,J ) , there is a canonical filtration-preserving chain isomorphism h(j,H ) : (CFk (H ), ∂(H,J ) ) → (CFk (H ), ∂(H,J ) ), where j is any homotopy from J and J , and H ≡ H is the constant homotopy of H . Therefore, from now on we suppress J -dependence on the Floer homology in our exposition unless it is absolutely necessary. For each given pair of real numbers λ, µ ∈ R \ Spec(H ) with λ < µ, we define (λ,µ]

CF∗

(H ) := CF µ (H )/CF λ (H ).

Then for each triple λ < µ < ν, where λ = −∞ or ν = ∞ are allowed, we have the short exact sequence of the complex of graded Q vector spaces (λ,µ]

0 → CFk

(λ,ν]

(H ) → CFk

(µ,ν]

(H ) → CFk

(H ) → 0

for each k ∈ Z. This then induces the long exact sequence of graded modules (λ,µ]

· · · → H Fk

(λ,ν]

(H ) → H Fk

(µ,ν]

(H ) → H Fk

(λ,µ]

(H ) → H Fk−1 (H ) → · · ·

whenever the relevant Floer homology groups are defined. We close this section by fixing our grading convention for H F∗ (H ). This convention is the analogue to the one used in [Oh1, Oh2] in the context of Lagrangian submanifolds. We first recall that solutions of the negative gradient flow equation of −f , (i.e., of the positive gradient flow of f χ˙ − grad f (χ ) = 0 corresponds to the negative gradient flow of the action functional Af ). This gives rise to the relation between the Morse indices µMorse −f (p) and the Conley–Zehnder =]; f ) (see [SZ, Lemma 7.2] but with some care about the different indices µCZ ([p, p convention of the Hamiltonian vector field. Their definition of XH is −XH in our convention):

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Y.-G. Oh

µCZ ([p, p =]; f ) = µMorse −f (p) − n

(4.14)

in our convention. On the other hand, obviously we have Morse (p)) − n = n − µMorse (p). µMorse −f (p) − n = (2n − µf f

We will always grade H F∗ (H ) by the Conley–Zehnder index k = µH ([z, w]) := µCZ ([z, w]; H ).

(4.15)

This grading convention makes the degree k of [q, = q ] in CFk (f ) coincides with the Morse index of q of f for each q ∈ Crit f . Recalling that we chose the Morse complex CM∗ (−f ) ⊗ ↓ for the quantum chain complex CQ∗ (−f ), it also coincides with the standard grading of the quantum cohomology via the map 0 : QH k (M) → QH2n−k (M). Form now on, we will denote by µH ([z, w]) the Conley–Zehnder index of [z, w] for the Hamiltonian H . Under this grading, we have the following grading-preserving isomorphism QH n−k (M) → QHn+k (M) ∼ = H Qn+k (−f ) → H Fk (f ) → H Fk (H ). (4.16) We will also show in Section 6 that this grading convention makes the pants product, denoted by ∗, having the degree −n: ∗ : H Fk (H ) ⊗ H F (K) → H F(k+)−n (H #K)

(4.17)

which will be compatible with the degree-preserving quantum product · : QH a (M) ⊗ QH b (M) → QH a+b (M).

5 Construction of the spectral invariants of Hamiltonian functions In this section, we associate some homologically essential critical values of the action functional AH to each Hamiltonian functions H and quantum cohomology class a, and call them the spectral invariants of H . We denote this assignment by ∞ ([0, 1] × M) × QH ∗ (M) → R ρ : Cm

as described in the introduction of this paper. Before launching our construction, some overview of our construction of spectral invariants is necessary. 5.1 Overview of the construction We recall the canonical isomorphism

Spectral invariants

545

hαβ : H F∗ (Hα ) → H F∗ (Hβ ) which satisfies the composition law hαγ = hαβ ◦ hβγ . We denote by H F∗ (M) the corresponding model Q-vector space. We also note that H F∗ (H ) is induced by the filtered chain complex (CF∗λ (H ), ∂), where CF∗λ (H ) = spanQ {α ∈ CF∗ (H ) | λH (α) ≤ λ}, i.e., the subcomplex generated by the critical points [z, w] ∈ Crit AH with AH ([z, w]) ≤ λ. Then there exists a canonical inclusion iλ : CF∗λ (H ) → CF∗∞ (H ) := CF∗ (H ) which induces a natural homomorphism iλ : H F∗λ (H ) → H F∗ (H ). For each given element ∈ F H∗ (M) and Hamiltonian H , we represent the class by a Novikov cycle α of H and measure its level λH (α), and define ρ(H ; ) := inf {λ ∈ R | ∈ Im iλ } or, equivalently, ρ(H ; ) :=

inf

α;iλ [α]=

λH (α).

The crucial task then is to prove that for each (homogeneous) element = 0, the value ρ(H ; ) is finite, i.e., “the cycle α is linked and cannot be pushed to infinity by the negative gradient flow of the action functional.’’ In the classical critical point theory (see [BnR], for example), this property of semiinfinite cycles is called the linking property. We like to point out that there is no manifest way to see the linking property or the critical nature of the mini-max value ρ(H ; ) from the definition itself. We will prove this finiteness first for the Hamiltonian f , where f is a Morse function and is sufficiently small. This finiteness strongly relies on the facts that the Floer boundary operator ∂f in this case has the form Morse ⊗ ω , ∂f = ∂−f

(5.1)

i.e., “there is no quantum contribution on the Floer boundary operator,’’ and the Morse cannot push down the level of a nontrivial classical Morse theory proves that ∂−f cycle more than − max f (see [Oh4]). Once we prove the finiteness for f , then we consider the general nondegenerate Hamiltonian H . We compare the cycles in CF∗ (H ) and the transferred cycles in CF∗ (f ) by the chain map h−1 H : CF∗ (H ) → CF∗ (f ), where H is a homotopy

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connecting f and H . The change of the level can then be measured by judicious use of (4.7) and Remark 4.5 which will prove the finiteness for any H . After we prove finiteness of ρ(H ; a) for general H , we study the continuity property of ρ(H ; a) under the change of H . This will be done, via the equation (4.6), considering the level change between arbitrary pair (H, K). Finally, we prove that the limit lim ρ(f ; )

→0

exists and is independent of the choice of Morse function f . If the Floer homology class is identified with a 0 for a quantum cohomology class a ∈ QH ∗ (M) under the PSS-isomorphism [PSS], then this limit is nothing but the valuation v(a). In this procedure, we can avoid considering the “singular limit’’ of the “chains.’’ (See [Oh8, Section 8] for some illustration of the difficulty in studying such limits.) We only need to consider the limit of the values ρ(H ; ) as H → 0 which is a much simpler task than considering the limit of chains which involves highly nontrivial analytical work. (We refer to the forthcoming work [FOh2] for the consideration of this limit in the chain level.) 5.2 Finiteness; the linking property of semiinfinite cycles With this overview, we now start with our construction. We first recall the natural pairing ·, · : CQ∗ (−f ) ⊗ CQ∗ (−f ) → Q, where we have CQk (−f ) := (CMk (−f ), ∂−f ) ⊗ ↓ , CQk (−f ) := (CM2n−k (f ), ∂f ) ⊗ ↑ .

Remark 5.1. We would like to emphasize that in our definition CQk (−f ) is not isomorphic to HomQ (CQk (−f ), Q) in general. However, there is a natural homomorphism CQk (−f ) → HomQ (CQk (−f ), Q); a → a, · (5.2) whose image lies in the subset of continuous linear functionals Homcont (CQk (−f ), Q) := CQkcont (−f ) ⊂ HomQ (CQk (−f ), Q). See the appendix for more discussions on this aspect. We would like to emphasize that (5.2) is well defined because of the choice of directions of the Novikov rings ↑ and ↓ . In general, the map (5.2) is injective but not an isomorphism. Polterovich [Po4, EnP] observed that this point is closely related to a certain failure of “Poincaré duality’’ of the Floer homology with Novikov rings as its coefficients.

Spectral invariants

547

Now we are ready to give the definition of our spectral invariants. Previously in [Oh4], the author outlined this construction for the classical cohomology class in H ∗ (M) ⊂ QH ∗ (M). Definition 5.2. Let H be a generic nondegenerate Hamiltonian. For each given a ∈ QH k (M) ∼ = H Qk (−f ), we define ρ(H, a) = inf {λH (α) | [α] = a 0 , α ∈ CFk (H )}. α

(5.3)

Theorem 5.3. Let 0 = a ∈ QH ∗ (M). (1) Let H be a generic nondegenerate Hamiltonian. Then ρ(H, a) is finite. (2) For any pair of generic nondegenerate Hamiltonians H, K, we have the inequality

1

1

− max(K − H )dt ≤ ρ(K, a) − ρ(H, a) ≤

0

− min(K − H )dt. (5.4)

0

0 ([0, 1]×M). In particular, the function H → ρ(H ; a) continuously extends to Cm

Proof. We will prove the finiteness in two steps: first we prove the finiteness for f for sufficiently small > 0 for any given Morse function f , and then we prove it for general H using this finiteness for f . After this we will prove the inequality (5.4). Step 1: The finiteness of for f . Let f be any fixed Morse function and fix > 0 so small that there is no quantum contribution for the Floer boundary operator ∂(f,J0 ) for a time independent family Jt ≡ J0 for any compatible almost complex structure J0 , i.e., we have Morse ∂(f,J0 ) ! ∂−f ⊗ ↓ω . (5.5) It is well known [Fl, FOn, LT1] that this is possible. Fixing such and J0 , we denote ∂f = ∂(f,J0 ) . Then by considering the Morse homology of −f with respect to the Riemannian metric gJ0 = ω(·, J0 ·), we have the identity Morse Morse QH ∗ (M) ∼ ⊗ ↑ / Im ∂f ⊗ ↑ = H M∗ (f ) ⊗ ↑ , = ker ∂f Morse Morse QH∗ (M) ∼ ⊗ ↓ / Im ∂−f ⊗ ↓ = H M∗ (−f ) ⊗ ↓ . = ker ∂−f

Recalling

CFk (f ) ∼ = CQn+k (−f ),

from (5.5), we represent a 0 ∈ QHn+k (M) by a Novikov cycle of f , where α= ap⊗q A p ⊗ q A A

with ap ∈ Q and p ∈ Crit ∗ (−f ) and

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Y.-G. Oh

n + k = µf (p ⊗ q A ),

(5.6)

where µf (p ⊗ q A ) is the Conley–Zehnder index of the element p ⊗ q A = [p, p =#A]. We recall the general index formula µH ([z, w ⊗ A]) = µH ([z, w]) + 2c1 (A) in our convention (see [Oh9] for the proof of this index formula). Applying this to H = f , we have obtained µf ([p, p =#A]) = µf ([p, p =]) + 2c1 (A). Combining this with µMorse =]) + n, −f (p) = µf ([p, p we derive that (5.6) is equivalent to µMorse −f (p) = n + k − 2c1 (A). Next, we see that α has the level λf (α) = max{−f (p) − ω(A) | ap⊗q A = 0}

(5.7)

because Af ([p, p =#A]) = −f (p) − ω(A). Now the most crucial point in our construction is to prove the finiteness inf λf (α) > −∞.

(5.8)

[α]=a 0

The following lemma proves this linking property. We first like to point out that the quantum cohomology class a= aA q −A A

uniquely determines the set (a) := {A ∈ | aA = 0}. By the finiteness condition in the formal power series, we can enumerate (a) so that λ1 > λ2 > λ3 > · · ·

(5.9)

without loss of generality. In particular, we have v(a) = −ω(A1 ) = λ1 .

(5.10)

Lemma 5.4. Let a = QH n−k (M) and a 0 ∈ QHn+k (M) its dual. Suppose that a0 = aj q Aj j

Spectral invariants

549

with 0 = aj ∈ Hn+k−2c1 (Aj ) (M), where λj = −ω(Aj ) are arranged as in (5.9). Denote by γ a Novikov cycle of f with [γ ] = a 0 ∈ H Fk (f ) ∼ = QHn+k (M) and define the gap c(a) := λ1 − λ2 . Then we have 1 1 v(a) − c(a) ≤ inf {λf (γ ) | [γ ] = a 0 } ≤ v(a) + c(a) γ 2 2

(5.11)

for any sufficiently small > 0 and, in particular, (5.8) holds. We also have lim inf {λf (γ ) | [γ ] = a 0 } = v(a)

→0 γ

(5.12)

and so the limit is independent of the choice of Morse functions f . Proof. We represent a 0 by a Novikov cycle γA q A , γj ∈ CM∗ (−f ) γ = A

of f . It follows from (5.3) that if A ∈ (a), all the coefficient Morse chains in this sum must be cycles, and if A ∈ / (a), the corresponding coefficient cycle must be a boundary. Therefore, we can decompose γ as γ = γ(a) + γ(a) C,

(5.13)

where γ(a) :=

γA q A ,

A∈(a)

γ(a) C :=

γB q B ,

B ∈(a) /

and we have γ(a) C = ∂f (ν) for some Floer chain ν of f . Since the summands in γ(a) C cannot cancel those in γ(a) , we have ⎛ ⎞ λf (γ ) ≥ λf (γ(a) ) = λf ⎝ γA q A ⎠ . A∈(a)

Therefore, by removing the exact term ∂f (ν) when we take the infimum over the cycles γ with [γ ] = a 0 for the definition of ρ(f ; a), we may always assume that γ has the form γ = γj q Aj j

550

Y.-G. Oh

with Aj ∈ (a). Then again by (5.5), we have [γj ] = aj ∈ H∗ (M). Furthermore, we note that we have −ω(Aj ) − max(f ) ≤ λf (γj q Aj ) ≤ −ω(Aj ) − min(f ). Therefore, if we choose > 0 so small that (max f − min f ) ≤ c(a) = λ1 − λ2 , then we have λf (γ1 q A1 ) ≥ λf (γj q Aj ) for all j = 1, 2, . . . , and so λf (γ ) = λf (γ1 q A1 ). Combining them, we derive −ω(A1 ) − max f ≤ λf (γ ) ≤ −ω(A1 ) + max f. (5.11) follows from (5.14) if we choose so that (max f − min f ) < also immediately follows from (5.14).

(5.14) c(a) 2 .

(5.12)

Step 2: The finiteness for general H . Now we consider generic nondegenerate H s. We fix f be any Morse function and and > 0 as in Lemma 5.4. Let α ∈ CF∗ (H ) be a Floer cycle of H with [α] = a 0 , and H = Hlin the linear homotopy Hlin : s → (1 − s)(f ) + sH. Applying (4.12) to the “inverse’’ linear homotopy −1 Hlin : s → (1 − s)H + s(f ),

we obtain the inequality λf (hH−1 (α)) ≤ λH (α) + lin

1

− min(f − H )dt.

(5.15)

0

More precisely, it follows from the definition of the chain map hH−1 that for any lin generator [z , w ] of the cycle hH−1 (α) of f , there is a generator [z, w] of the cycle lin α such that the equation (4.6) has a solution. Then we derive, from (4.11), 1 Af ([z , w ]) ≤ AH ([z, w]) + − min (f − Ht )dt 0

1

≤ λH (α) + 0

x∈M

− min (f − Ht )dt. x∈M

Spectral invariants

551

−1 Since this holds for any generator [z , w ] of Hlin (α), we obtain

−1 λf (Hlin (α)) ≤ λH (α) +

1 0

− min (f − Ht )dt. x∈M

(5.16)

−1 (α)] = a 0 that we have On the other hand, it follows from [Hlin −1 ρ(a; f ) ≤ λf (Hlin (α)).

Combining this with (5.16), we derive '

1

λH (α) ≥ ρ(a; f ) −

* − min (f − Ht )dt . x∈M

0

(5.17)

Since this holds for any cycle α of H with [α] = a 0 , by taking the infimum over all such α in (5.17), we have finally obtained ' * 1

ρ(H ; a) ≥ ρ(a; f ) − 0

− min (f − Ht )dt . x∈M

(5.18)

Since Lemma 5.4 shows that ρ(a; f ) > −∞, this implies in particular that ρ(H ; a) > −∞ and so ρ(H ; a) is finite. Step 3: Proof of (5.4). Finally, we prove the inequality (5.4). For this purpose, we consider general generic nondegenerate pairs H, K. Let δ > 0 be any given number. We choose a cycle α of H , respectively, so that [α] = a 0 and λH (α) ≤ ρ(H ; a) + δ.

(5.19)

We would like to emphasize that this is possible, because we have already shown that ρ(H ; a) > −∞. By considering the linear homotopy hlin H K from H to K, we derive λK (hlin − min(Kt − Ht )dt. (5.20) H K (α)) ≤ λH (α) + x

On the other hand (5.19) implies that λH (α) + − min(Kt − Ht )dt x ≤ ρ(H ; a) + δ + − min(Kt − Ht )dt.

(5.21)

x

0 Since [hlin H K (α)] = a , we have

λK (hlin H K (α)) ≥ ρ(K; a) by the definition of ρ(K; a). Combining (5.20)–(5.22), we have derived

(5.22)

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Y.-G. Oh

1

ρ(K; a) − ρ(H ; a) ≤ δ +

− min(Kt − Ht )dt. x

0

Since this holds for arbitrary δ, we have derived 1 ρ(K; a) − ρ(H ; a) ≤ − min(Kt − Ht )dt. 0

x

By changing the role of H and K, we also derive 1 ρ(H ; a) − ρ(K; a) ≤ − min(Ht − Kt )dt = 0

x

1 0

Hence we have the inequality 1 − max(Kt − Ht )dt ≤ ρ(K; a) − ρ(H ; a) ≤ 0

x

1 0

max(Kt − Ht )dt. x

− min(Kt − Ht )dt x

which is precisely (5.4). Obviously the inequality (5.4) enables us to extend the definition of ρ by continuity to arbitrary C 0 -Hamiltonians. This finishes the proof of Theorem 5.3.

6 Basic properties of the spectral invariants In this section, we will prove all the remaining properties stated in Theorem I in the introduction. We first restate the main axioms of the spectral invariants. Theorem 6.1. Let H, F be arbitrary smooth Hamiltonian functions, and a = 0 ∈ QH ∗ (M) and let ∞ ρ : Cm ([0, 1] × M) × QH ∗ (M) → R be as defined in Section 5. Then ρ satisfies the following properties: (1) Projective invariance: ρ(H ; λa) = ρ(H ; a) for any 0 = λ ∈ Q. (2) Normalization: For a = A∈ aA ⊗ q A , ρ(0; a) = v(a), the valuation of a. ; a) for any symplectic diffeomor(3) Symplectic invariance: ρ(η∗ H ; a) = ρ(H phism η. (4) Triangle inequality: ρ(H #F ; a · b) ≤ ρ(H ; a) + ρ(F ; b). (5) C 0 -continuity: |ρ(H ; a) − ρ(F ; a)| ≤ H ◦ F = H − F and, in particular, ρ(·, a) is continuous with respect to the C 0 -topology of Hamiltonian functions. We have already proved the properties of normalization and C 0 -continuity in the course of proving the linking property of the Novikov Floer cycles in Section 5. The remaining parts of the proofs deal with the symplectic invariance and the triangle inequality. 6.1 Proof of symplectic invariance We consider the symplectic conjugation

Spectral invariants

φ → η−1 φη;

553

Ham(M, ω) → Ham(M, ω)

for any symplectic diffeomorphism η : (M, ω) → (M, ω). Recall that the pullback function η∗ H given by η∗ H (t, x) = H (t, η(x)) (6.1) generates the conjugation η−1 φη when H → φ. We summarize the basic facts on this conjugation relevant to the filtered Floer homology here: (1) (2) (3) (4)

When H → φ, η∗ H → ηφη−1 . If H is nondegenerate, η∗ H is also nondegenerate. If (J, H ) is regular in the Floer-theoretic sense, then so is (η∗ J, η∗ H ). There exists natural bijection η∗ : 0 (M) → 0 (M) defined by η∗ ([z, w]) = ([η ◦ z, η ◦ w]) under which we have the identity AH ([z, w]) = Aη∗ H (η∗ [z, w]).

(6.2)

(5) The L2 -gradients of the corresponding action functionals satisfy η∗ (grad J AH )([z, w]) = grad η∗ J (Aη∗ H )(η∗ ([z, w])).

(6.3)

(6) If u : R × S 1 → M is a solution of the perturbed Cauchy–Riemann equation for (J, H ), then η∗ u = η ◦ u is a solution for the pair (η∗ J, η∗ H ). In addition, all the Fredholm properties of (J, H, u) and (η∗ J, η∗ H, η∗ u) are the same. These facts imply that the conjugation by η induces the canonical filtration-preserving chain isomorphism η∗ : (CF∗λ (H ), ∂(H,J ) ) → (CF∗λ (η∗ H ), ∂(η∗ H,η∗ J ) ) for any λ ∈ R \ Spec(H ) = R \ Spec(η∗ H ). In particular, it induces a filtrationpreserving isomorphism η∗ : H F∗λ (H, J ) → H F∗λ (η∗ H, η∗ J ) in homology. The symplectic invariance is then an immediate consequence of our construction of ρ(H ; a). 6.2 Proof of the triangle inequality To start with the proof of the triangle inequality, we need to recall the definition of the “pants product’’ H F∗ (H ) ⊗ H F∗ (F ) → H F∗ (H #F ).

(6.4)

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Y.-G. Oh

We also need to straighten out the grading problem of the pants product. For the purpose of studying the effect on the filtration under the product, we need to define this product in the chain level in an optimal way as in [Oh2, Sc, En1]. For this purpose, we will mostly follow the description provided by Entov [En1] with few notational changes and a different convention on the grading. As pointed out before, our grading convention satisfies the relation (4.17) under the pants product. Except for the grading convention, the conventions in [En1, En2] for the definition of Hamiltonian vector field and the action functional coincide with our conventions in [Oh1, Oh2, Oh3, Oh5] and in this paper. Let be the compact Riemann surface of genus 0 with three punctures. We fix a holomorphic identification of a neighborhood of each puncture with either [0, ∞)×S 1 or (−∞, 0]×S 1 with the standard complex structure on the cylinder. We call punctures of the first type negative and the second type positive. In terms of the “pair of pants’’ \ ∪i Di , the positive puncture corresponds to the outgoing ends and the negative corresponds to the incoming ends. We denote the neighborhoods of the three punctures by Di , i = 1, 2, 3, and the identification by ϕi+ : Di → (−∞, 0] × S 1 for positive punctures and ϕ3− : D3 → [0, ∞) × S 1 for negative punctures. We denote by (τ, t) the standard cylindrical coordinates on the cylinders. We fix a cutoff function ρ + : (−∞, 0] → [0, 1] defined by + 1, τ ≤ −2, ρ= 0, τ ≥ −1 and ρ − : [0, ∞) → [0, 1] by ρ − (τ ) = ρ + (−τ ). We will just denote by ρ these cutoff functions for both cases when there is no danger of confusion. We now consider the (topologically) trivial bundle P → with fiber isomorphic to (M, ω) and fix a trivialization i : Pi := P |Di → Di × M on each Di . On each Pi , we consider the closed two-form of the type ωPi := ∗i (ω + d(ρHt dt))

(6.5)

for a time periodic Hamiltonian H : [0, 1] × M → R. The following is an important lemma whose proof we omit (see [En1]). Lemma 6.2. Consider three normalized Hamiltonians Hi , i = 1, 2, 3. Then there exists a closed two-form ωP such that (1) ωP |Pi = ωPi ;

Spectral invariants

555

(2) ωP restricts to ω in each fiber; (3) ωPn+1 = 0. Such ωP induces a canonical symplectic connection ∇ = ∇ωP [GLS, En1]. In addition it also fixes a natural deformation class of symplectic forms on P obtained by those

P ,λ := ωP + λω , where ω is an area form and λ > 0 is a sufficiently large constant. We will always normalize ω so that ω = 1. Next, let J be an almost complex structure on P such that (1) J is ωP -compatible on each fiber and so preserves the vertical tangent space; (2) the projection π : P → is pseudoholomorphic, i.e., dπ ◦ J = j ◦ dπ. When we are given three t-periodic Hamiltonian H = (H1 , H2 , H3 ), we say that J is (H, J )-compatible if J additionally satisfies (3) For each i, (i )∗ J = j ⊕ JHi , where t ∗ JHi (τ, t, x) = (φH ) J i

for some t-periodic family of almost complex structure J = {Jt }0≤t≤1 on M over a disc Di ⊂ Di in terms of the cylindrical coordinates. Here Di = ϕi−1 ((−∞, −Ki ] × S 1 ), i = 1, 2, and ϕ3−1 ([K3 , ∞) × S 1 ) for some Ki > 0. Later we will particularly consider the case where J is in the special form adapted to the Hamiltonian H . See (6.23). Condition (3) implies that the J-holomorphic sections v over Di are precisely the solutions of the equation ∂u ∂u + Jt − XHi (u) = 0 (6.6) ∂τ ∂t if we write v(τ, t) = (τ, t, u(τ, t)) in the trivialization with respect to the cylindrical coordinates (τ, t) on Di induced by φi± above. Now we are ready to define the moduli space which will be relevant to the definition of the pants product that we need to use. To simplify the notation, we denote = z = [z, w] in general and = z = (= z1 ,= z2 ,= z3 ), where = zi = [zi , wi ] ∈ Crit AHi for i = 1, 2, 3. Definition 6.3. Consider the Hamiltonians H = {Hi }1≤i≤3 with H3 = H1 #H2 , and let J be a H -compatible almost complex structure. We denote by M(H, J;= z) the space of all J-holomorphic sections u : → P that satisfy the following: (1) The maps ui := u ◦ (φi−1 ) : (−∞, Ki ] × S 1 → M, which are solutions of (6.6), satisfy lim ui (τ, ·) = zi , i = 1, 2, τ →−∞

and similarly for i = 3 changing −∞ to +∞.

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Y.-G. Oh

(2) The closed surface obtained by capping off prM ◦ u() with the discs wi taken with the same orientation for i = 1, 2, and the opposite one for i = 3 represents zero in π2 (M). Note that M(H, J;= z) depends only on the equivalence class of = zs: we say that = z ∼ = z if they satisfy zi = zi , wi = wi #Ai for Ai ∈ π2 (M) and 3i=1 Ai represents zero (mod) Z-torsion elements. The (virtual) dimension of M(H, J;= z) is given by dim M(H, J;= z) = 2n − (−µH1 (z1 ) + n) − (−µH2 (z2 ) + n) − (µH3 (z3 ) + n) = −n + (−µH3 (z3 ) + µH1 (z1 ) + µH2 (z2 )). (6.7) Note that when dim M(H, J;= z) = 0, we have n = −µH3 (= z3 ) + µH1 (= z1 ) + µH2 (= z2 ) which is equivalent to µH3 (= z3 ) = (µH1 (= z1 ) + µH2 (= z2 )) − n,

(6.8)

which provides the degree of the pants product (4.17) in our convention of the grading of the Floer complex we adopt in this paper. Now the pair-of-pants product ∗ for the chains is defined by = z1 ∗= z2 = #(M(H, J;= z))= z3 (6.9) = z3

for the generators = zi and then by linearly extending over the chains in CF∗ (H1 ) ⊗ CF∗ (H2 ). Our grading convention makes this product of degree −n. Now with this preparation, we are ready to prove the triangle inequality. Proof of the triangle inequality. Let α ∈ CF∗ (H ) and β ∈ CF∗ (F ) be Floer cycles with [α] = [β] = a 0 and consider their pants product cycle α ∗β := γ ∈ CF∗ (H #F ). Then we have [α ∗ β] = (a · b)0 and so ρ(H #F ; a · b) ≤ λH #F (α ∗ β).

(6.10)

Let δ > 0 be any given number and choose α ∈ CF∗ (H ) and β ∈ CF∗ (F ) so that δ 2 δ λH (β) ≤ ρ(F ; b) + . 2 λH (α) ≤ ρ(H ; a) +

Then we have the expressions

(6.11)

Spectral invariants

α=

ai [zi , wi ] with AH ([zi , wi ]) ≤ ρ(H ; a) +

i

557

δ 2

and β=

j

δ aj [zj , wj ] with AH ([zj , wj ]) ≤ ρ(H ; b) + . 2

Now using the pants product (6.9), we would like to estimate the level of the chain α#β ∈ CF∗ (H #F ). The following is a crucial lemma whose proof we omit, but we refer to [Sc, Section 4.1] or [En1, Section 5]. Lemma 6.4. Suppose that M(H, J;= z) is nonempty. Then we have the identity v ∗ ωP = −AH1 #H2 ([z3 , w3 ]) + AH1 ([z1 , w1 ]) + AH2 ([z2 , w2 ]) (6.12) for any ∈ M(H, J;= z). Now since v is J-holomorphic and J is P ,λ -compatible, we have ∗ ∗ ∗ 0 ≤ v P ,λ = v ωP + λ v ω = v ∗ ωP + λ. Lemma 6.5 ([En1, Theorems 3.6.1 and 3.7.4]). Let Hi s be as in Lemma 6.2. Then for any given δ > 0, we can choose a closed two-form ωP so that P ,λ = ωP + λω becomes a symplectic form for all λ ≥ δ. In other words, the size size(H ) (see [En1, Definition 3.1]) is ∞. We recall that from the definition of ∗ that for any [z3 , w3 ] ∈ α ∗ β there exist [z1 , w1 ] ∈ α and [z2 , w2 ] ∈ β such that M(J, H ;= z) is nonempty with the asymptotic condition = z = ([z1 , w1 ], [z2 , w2 ]; [z3 , w3 ]). Applying this and the above two lemmas to H and F for λ arbitrarily close to 0, and also applying (6.10) and (6.11), we immediately derive AH #F ([z3 , w3 ]) ≤ AH ([z1 , w1 ]) + AF ([z2 , w2 ]) + δ ≤ λH (α) + λF (β) + δ ≤ ρ(H ; a) + ρ(F ; b) + 2δ

(6.13)

for any [z3 , w3 ] ∈ α ∗ β. Combining (6.10), (6.11), and (6.13), we derive ρ(H #F ; a · b) ≤ ρ(H ; a) + ρ(F ; b) + 2δ. Since this holds for any δ, we have proved ρ(H #F ; a · b) ≤ ρ(H ; a) + ρ(F ; b). The triangle inequality mentioned in Theorem 6.1 immediately follows from the ; a) = ρ(H ; a) in Theorem 5.5. definition ρ(φ

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7 The rational case; proof of the spectrality In this section, we will prove the spectrality for the rational symplectic manifolds: we recall that a symplectic manifold (M, ω) is rational if the period group ω is discrete. We will further study the spectrality property on general symplectic manifolds elsewhere, which turns out to be much more nontrivial to prove. Theorem 7.1. Suppose that (M, ω) is rational. Then for any smooth one-periodic Hamiltonian function H : S 1 × M → R, we have ρ(H ; a) ∈ Spec(H ) for each given quantum cohomology class 0 = a ∈ QH ∗ (M). Proof. We need to show that the mini-max value ρ(H ; a) is a critical value, i.e., that 0 (M) such that there exists [z, w] ∈ AH ([z, w]) = ρ(H ; a), dAH ([z, w]) = 0, i.e.,

z˙ = XH (z).

(7.1)

We have already shown the finiteness of the value ρ(H ; a) in Section 5. If H is nondegenerate, we use the fixed Hamiltonian. If H is not nondegenerate, we approximate H by a sequence of nondegenerate Hamiltonians Hj in the C 2 topology. Let [zj , wj ] ∈ Crit AHj be the peak of a Floer cycle αj ∈ CF∗ (Hj ) such that lim AHj ([zj , wj ]) = ρ(H ; a).

j →∞

(7.2)

Such a sequence can be chosen from the definition of ρ(·; a) and the finiteness thereof. Since M is compact and Hj → H in the C 2 topology, and z˙ j = XHj (zj ) for all j , it follows from the standard bootstrap argument that zj has a subsequence, which we still denote by zj , converging to z∞ which solves z˙ = XH (z). Now we show 0 (M). Since we fix the quantum cohomology class that [zj , wj ] are precompact on 0 = a ∈ QH ∗ (M) (or more specifically since we fix its degree) and the Floer cycle satisfies [αj ] = a, we have µHj ([zj , wj ]) = µHi ([zi , wi ]).

(7.3)

0 (M) is a closed subset of R Lemma 7.2. When (M, ω) is rational, Crit(AK ) ⊂ for any smooth Hamiltonian K, and is locally compact in the subspace topology of the covering space 0 (M) → 0 (M). π : Proof. First note that when (M, ω) is rational, the covering group ω of π above is discrete. Together with the fact that the set of solutions of z˙ = XK (z) is compact (on compact M), it follows that 0 (M) | z˙ = XK (z)} Crit(AK ) = {[z, w] ∈ is a closed subset which is also locally compact.

Spectral invariants

559

Now consider the bounding discs of z∞ wj = wj #ucan j for all sufficiently large j , where ucan is the homotopically unique thin cylinder between zj and z∞ : more precisely, ucan j is given by the formula ξj (t) = (expzj (t) )−1 (z∞ (t)),

ucan j (s, t) = expzj (t) (sξj (t)),

(7.4)

where exp is the exponential map with respect to a fixed metric gJref = ω(·, Jref ·) for a fixed compatible almost complex structure. We note that as j → ∞ the geometric area of ucan j converges to 0. We compute the action of the critical points [z∞ , wj ] ∈ Crit AH , AH ([z∞ , wj ])

=−

wj

ω−

=−

1

ω−

wj

' = −

0

ucan j

0

H (t, z∞ (t))dt *

Hj (t, zj (t))dt 0

1

−

1

ω−

1

ω−

wj

'

(7.5)

H (t, z∞ (t))dt

0

H (t, z∞ (t)) − '

= AHj ([zj , wj ]) −

1 0

1

*

Hj (t, zj (t)) −

0

H (t, z∞ (t)) −

1

ω ucan j

*

Hj (t, zj (t)) −

0

From the explicit expression (7.4), it follows that ω=0 lim j →∞ ucan j

ω. ucan j

(7.6)

since the geometric area of ucan j converges to zero, and we have can Area(uj ) ≥ ω . ucan j

Since zj converges to z∞ uniformly and Hj → H , we have ' * 1

− 0

H (t, z∞ (t)) −

1

H (t, zj (t)) → 0.

0

Therefore, combining (7.2), (7.6), and (7.7), we derive lim AH ([z∞ , wj ]) = ρ(H ; a).

j →∞

(7.7)

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Y.-G. Oh

In particular, AH ([z∞ , wj ]) is a Cauchy sequence, which implies that ω− w w j

i

ω = AH ([z∞ , wj ]) − AH ([z∞ , wi ]) → 0;

i.e.,

Since ω is discrete and

wj #w i

wj #w i

ω → 0.

ω ∈ ω , this indeed implies that wj #w i

ω=0

(7.8)

for all sufficiently large i, j . Since the set { w ω}j ∈Z+ ⊂ R is bounded, these imply j that the sequence w ω eventually stabilizes. Going back to (7.5), we have proved j

that the actions

AH ([z∞ , wj ])

stabilize, and so we have AH ([z∞ , wN ]) = lim AH ([z∞ , wj ]) = ρ(H ; a) j →∞

for a fixed sufficiently large N ∈ Z+ . This proves that ρ(H ; a) is indeed a critical ]. This finishes the proof. value of AH at the critical point [z∞ , wN

We now state the following theorem. ∞ (M × [0, 1], R) the set of normalized Theorem 7.3. Let (M, ω) be rational and Cm ∞ ∞ (M × [0, 1], R) → R the extended C -Hamiltonians on M. We denote by ρa : Cm continuous function defined by ρa (H ) = ρ(H ; a).

= [φ, H ]. Hence ρa (1) The image of ρa depends only on the homotopy class φ pushes down to a well-defined function ρ : Ham(M, ω) × QH ∗ (M) → R;

; a) := ρ(H ; a) ρ(φ

(7.9)

= [φ, H ]. for any H with φ (2) We have the formula ρ(H ; a) = inf {λ | a 0 ∈ Im(iλ : H F∗λ (H ) → H F∗ (H ))}. λ

(7.10)

Proof. We have shown in Theorem 7.1 that ρ(H ; a) is indeed a critical value of AH , i.e., lies in Spec(H ). With this fact, the well-definedness of the definition (7.9), i.e., = [φ, H ] is an immediate consequence of the combination independence of H with φ of the following results:

Spectral invariants

561

(1) H → ρ(H ; a) is continuous. (2) Spec(H ) is a measure zero subset of R (Lemma 2.2). ) depends only on its homotopy class [H ] = φ and so fixed (3) Spec(H ) = Spec(φ as long as [H ] = φ (Theorem 2.3). (4) The only real-valued continuous function from a connect space (e.g., the unit interval [0, 1]) whose image has measure zero in R is a constant function. (7.10) is just a rephrasing of the definition of ρ(H ; a). This finishes the proof of Theorem 7.3.

One more important property concerns the effect of ρ under the action of π0 (G). ∗ acts on Ham(M, ω) × QH (M) following (and adapting We first explain how π0 (G) into cohomological version) Seidel’s description of the action on QH∗ (M).According acts on QH∗ (M) by the quantum product of an to [Se], each element [h, h] ∈ π0 (G) even element #([h, h]) on QH∗ (M). We take the adjoint action of it on a ∈ QH ∗ (M) and denote it by h∗ a. More precisely, h∗ a is defined by the identity h∗ a, β = a, #([h, h]) · β

(7.11)

with respect to the nondegenerate pairing ·, · between QH ∗ (M) and QH∗ (M). act on Ham(M, Theorem 7.4 (monodromy shift). Let π0 (G) ω) × QH ∗ (M) as above, i.e., , a) = (h · φ , [h, h] · (φ h∗ a). (7.12) Then we have

; a)) = ρ(φ ; a) + Iω ([h, h]). ρ([h, h] · (φ

Proof. This is immediate from the construction of #([h, h]) in [Se]. Indeed, the map [h, h]∗ : CF∗ (F ) → CF∗ (H #F ) is induced by the map and we have

(7.13)

[z, w] → h([z, w]),

AH #F ( h([z, w])) = AF ([z, w]) + Iω ([h, h])

by (2.5). Furthermore, the map (7.12) is a chain isomorphism whose inverse is given by ([h, h]−1 )∗ . This immediately implies the theorem from the construction of ρ. Remark 7.5. Strictly speaking, h∗ a may not lie in the standard quantum cohomology ∗ QH (M) because it is defined as the linear functional on the complex CQ∗ (M) that is dual to the Seidel element #([h, h]) ∈ CQ∗ (M) under the canonical pairing between CQ∗ (M) and CQ∗ (M). A priori, the bounded linear functional h∗ a = #([h, h]), · may not lie in the image of : QH∗ (M) → QH ∗ (M), mentioned in Section 3, in general. In that case, one should consider h∗ a as a continuous quantum cohomology

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Y.-G. Oh

class in the sense of the appendix. We refer readers to the appendix for the explanation on how to extend the definition of our spectral invariants to the continuous quantum cohomology classes. Now we can define ρ : Ham(M, ω) × QH ∗ (M) by putting

; a) := ρ(H ; a) ρ(φ

with [H ] = φ when φ is nondegenerate, and then extending to for any H → φ arbitrary φ by continuity. ; a) for each a ∈ QH ∗ (M), we have constructed Then by the spectrality of ρ(φ continuous “sections’’ of the action spectrum bundle Spec(M, ω) → Ham(M, ω). by We define the essential spectrum of φ ) := {ρ(φ ; a) | 0 = a ∈ QH ∗ (M)}, spec(φ ) := {ρ(φ ; a) | 0 = a ∈ QH k (M)} speck (φ and the bundle of essential spectra by spec(M, ω) =

A

); spec(φ

∈H φ am(M,ω)

similarly for speck (M, ω).

8 Remarks on transversality Our construction of various maps in the Floer homology works as in the previous section for the strongly semipositive case [Se, En1] by the standard transversality argument. On the other hand, in the general case where constructions of operations in the Floer homology theory require the machinery of virtual fundamental chains through multivalued abstract perturbation [FOn, LT1, Ru], we need to explain how this general machinery can be incorporated into our construction. The full details will be provided elsewhere. We will use the terminology “Kuranishi structure’’ adopted by Fukaya and Ono [FOn] for the rest of the discussion. One essential point in our proofs is that various numerical estimates concerning the critical values of the action functional and the levels of relevant Novikov cycles do not require transversality of the solutions of the relevant pseudoholomorphic sections, but depends only on the nonemptiness of the moduli space M(H, J;= z)

Spectral invariants

563

which can be studied for any, not necessarily generic, Hamiltonian H . Since we always have suitable a priori energy bound which requires some necessary homotopy assumption on the pseudoholomorphic sections, we can compactify the corresponding moduli space into a compact Hausdorff space, using a variation of the notion of stable maps in the case of nondegenerate Hamiltonians H . We denote this compactification again by M(H, J;= z). This space could be pathological in general. But because we assume that the Hamiltonians H are nondegenerate, i.e., all the periodic orbits are nondegenerate, the moduli space is not completely pathological but at least carries a Kuranishi structure in the sense of Fukaya–Ono [FOn] for any H -compatible J. This enables us to apply the abstract multivalued perturbation theory and to perturb the compactified moduli space by a Kuranishi map + so that the perturbed moduli space M(H, J;= z, +) is transversal in that the linearized equation of the perturbed equation ∂ J(v) + +(v) = 0 is surjective and so its solution set carries a smooth (orbifold) structure. Furthermore, the perturbation + can be chosen so that as + → 0, the perturbed moduli space M(H, J;= z, +) converges to M(H, J;= z) in a suitable sense (see [FOn] for the precise description of this convergence). Now the crucial point is that nonemptiness of the perturbed moduli space will be guaranteed as long as certain topological conditions are met. For example, the followings are the prototypes that we have used in this paper: (1) hH1 : CF0 (f ) → CF0 (H ) is an isomorphism in homology and so [hH1 (10 )] = 0. This is immediately translated as an existence result of solutions of the perturbed Cauchy–Riemann equation. (2) The definition of the pants product ∗ and the identity [α ∗ β] = (a · b)0 in homology guarantee nonemptiness of the relevant perturbed moduli space M(H, J;= z, +) for α ∈ CF∗ (H1 ), β ∈ CF∗ (H2 ) with [α] = a 0 , and [β] = b0 , respectively. Once we prove the nonemptiness of M(H, J;= z, +) and an a priori energy bound for the nonempty perturbed moduli space and if the asymptotic conditions= z are fixed, we can study the convergence of a sequence vj ∈ M(H, J;= z, +j ) as +j → 0 by the Gromov–Floer compactness theorem. However, a priori there are infinite possibilities of asymptotic conditions for the pseudoholomorphic sections that we are studying, because we typically impose that the asymptotic limit lie in certain Novikov cycles like = z1 ∈ α,

= z2 ∈ β,

= z3 ∈ α ∗ β.

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Y.-G. Oh

Because the Novikov Floer cycles are generated by an infinite number of critical points [z, w] in general, one needs to control the asymptotic behavior to carry out the compactness argument. For this purpose, we need to establish a lower bound for the actions which will enable us to consider only finite possibilities for the asymptotic conditions because of the finiteness condition in the definition of Novikov chains. We would like to emphasize that obtaining a lower bound is the heart of the matter in the classical mini-max theory of the indefinite action functional which requires a linking property of semiinfinite cycles. On the other hand, obtaining an upper bound is usually an immediate consequence of the identity as in (4.10). With such a lower bound for the actions, we may then assume, by taking a subsequence if necessary, that the asymptotic conditions are fixed when we take the limit and so we can safely apply the Gromov–Floer compactness theorem to produce a (cusp)-limit lying in the compactified moduli space M(H, J;= z). This will then justify all the statements and proofs in the previous sections for the complete generality.

Appendix: Continuous quantum cohomology In this appendix, we define the genuinely cohomological version of the quantum cohomology and explain how we can extend the definition of the spectral invariants to the classes in this cohomological version. We call this continuous quantum cohomology and denote it by ∗ QHcont (M).

In this respect, we call the usual quantum cohomology ring QH ∗ (M) = H ∗ (M) ⊗ ∗ (M) and QH ∗ (M) ↑ the finite quantum cohomology. We call elements in QHcont continuous (respectively, finite) quantum cohomology classes. ∗ (M). Let f be a Morse We first define the chain complex associated to QHcont function and consider the complex of Novikov chains CQ2n−k (−f ) = CM2n−k (−f ) ⊗ ↓ (= CFk (f )).

(A.1)

On nonexact symplectic manifolds, this is typically infinite dimensional as a Q-vector space. Therefore, it is natural to put some topology on it rather than to consider it only as an algebraic vector space. For this purpose, we recall the definition of the level λ(α) = λf (α) of an element: α= αA q A , αA ∈ CM∗ (−f ): A

λ(α) = max{Af (αA q A ) | αA = 0} = max{λMorse −f (αA ) − ω(A)}. As we saw before, this level function satisfies the inequality λ(α + β) ≤ max{λ(α), λ(β)}

(A.2)

Spectral invariants

565

and provides a natural filtration on CQ2n−k (−f ), which defines a non-Archimedean topology. We refer to [Br] for a nice exposition to the non-Archimedean topology and geometry. Definition and Proposition A.1. For each degree ∗, consider the collection A B= {U (α, R) ⊂ CQ∗ (−f )} α∈CQ∗ (−f ),R∈R

of the subsets U (α, R) defined by U (α, R) = {β ∈ CQ∗ (−f ) | λ(β − α) < R}. Then B satisfies the properties of a basis of topology. We equip CQ∗ (−f ) with the topology generated by the basis B. Proof. We need to prove that for any given U (α1 , R1 ) and U (α2 , R2 ) with U (α1 , R1 )∩ U (α2 , R2 ) = ∅ and for any β ∈ U (α1 , R1 ) ∩ U (α2 , R2 ), there exists R3 such that U (α, R3 ) ⊂ U (α1 , R1 ) ∩ U (α2 , R2 ).

(A.3)

Let β ∈ U (α1 , R1 ) ∩ U (α2 , R2 ). Then β satisfies λ(β − αi ) < Ri ,

i = 1, 2.

(A.4)

Suppose γ ∈ U (β, R), where R is to be determined. Then we derive from (A.2) λ(γ − αi ) ≤ max{λ(γ − β), λ(β − αi )} = max{R, Ri }.

(A.5)

Therefore, if we choose R ≤ min{R1 , R2 }, then we will have U (β, R) ⊂ U (α1 , R1 ) ∩ U (α2 , R2 ), which finishes the proof of the fact that B really defines a basis of topology.

By the non-Archimedean triangle inequality (A.2), it follows that the basis element U (α, R) is nothing but the affine subspace R U (α, R) = CQR ∗ (−f ) + α = CF2n−∗ (f ) + α,

where CF∗R is defined as in Section 4. The following is an easy consequence of the definition of the boundary operator. Lemma A.2. The boundary operator Morse ∂f = ∂−f ⊗ : CQ2n−k (−f ) → CQ2n−k−1 (−f )

is continuous with respect to this topology. Proof. Let U (α, R) be a basis element and consider the preimage

566

Y.-G. Oh

(∂f )−1 (U (α, R)). Suppose β ∈ (∂f )−1 (U (α, R)), i.e., ∂f (β) ∈ U (α, R) and so λ(∂f (β) − α) < R.

(A.6)

λ(∂f (δ)) ≤ λ(δ)

(A.7)

Recall that for any Novikov Floer chain δ. Now we consider the basis element U (β, R). Then if γ ∈ U (β, R), we have λ(∂f (γ ) − α) ≤ max{λ(∂f (γ − β)), λ(∂f (β) − α)} ≤ max{λ(γ − β), λ(∂f (β) − α)}

(A.8)

< max{R, R} = R, where the second inequality comes from (A.7). This finishes the proof of ∂f (U (β, R)) ⊂ U (α, R), i.e., U (β, R) ⊂ (∂f )−1 (U (α, R) for any β ∈ U (α, R). Hence the proof.

Now we define the following. Definition A.3. A linear functional µ : CQ2n−k (−f ) → Q is called continuous (or bounded) if it is continuous with respect to the topology induced by the above filtration. We denote by CQcont (−f ) the set of continuous linear functionals on CQ2n−k (−f ). The following is easy to see from the definition of Novikov chains. Lemma A.4. A linear functional µ is continuous if and only if there exists λµ ∈ R such that µ(αA q A ) = 0 (A.9) for all A with −ω(A) ≤ λµ . Proof. The sufficiency part of the proof is easy and so we will focus on the necessary condition. We will prove this by contradiction. Suppose that µ : CQ2n−k (−f ) → Q is a continuous linear functional, but there exists a sequence of Aj with −ω(Aj ) → −∞,

i.e.,

ω(Aj ) → +∞

(A.10)

and αj ∈ CM∗ (−f ) such that µ(αj q Aj ) = 0. Now consider the sequence of Novikov chains

(A.11)

Spectral invariants

βN =

N

αj q Aj .

567

(A.12)

j =1

It is easy to check from (A.10) that βN converges to the Novikov chain β=

∞

αj q Aj

j =1

in the given non-Archimedean topology on CQ∗ (−f ). In fact, this convergence holds for the sequence N βc,N = (cj αj )q Aj (A.13) j =1

for any given sequence c = {cj ∈ Q}1≤j 3 is 0.

(An alternate nomenclature would refer to such an algebra as an L3 -algebra.) Of course, many of these 0s follow just from the fact that Xn = 0 for n ≥ 1, in contrast to the L∞ -structures that appear in the work of Fulp, Lada, and myself concerning higher spin algebras [FLS02b, FLS02a] where the complex is of the form X0 → X 1 (see Section 6.2 below).

5 Homological reduction of constrained Poisson algebras Cohomological physics had a major breakthrough with the “ghosts’’ introduced by Fade’ev and Popov [FP67]. These were incorporated into what came to be known as BRST cohomology (Becchi–Rouet–Stora [BRS75] and Tytutin [Tyu75]) and which was applied to a variety of problems in mathematical physics. There the ghosts were reinterpreted by Stora [Sto77] and others in terms of the Maurer–Cartan forms in the case of a finite-dimensional Lie group and more generally as generators of the Chevalley–Eilenberg cochain complex [CE48] for Lie algebra cohomology. If, as geometers, you feel more comfortable with manifolds, one can make the following algebra seem more palatable as functions on “supermanifolds,’’ but most (all?) of the work is just algebraic (homological). Warning! The term “BRST cohomology’’ has a variety of meanings in the existing literature. From time to time, it threatens to be used for any cohomology in physics, at least if the coboundary operator is called “Q.’’At other times, it refers (only implicitly) to the case in which the Lie algebra is the Virasoro algebra. I prefer to reserve the term for situations in which the coboundary operator has at least some part corresponding to that of Chevalley–Eilenberg. Such is the case for the ghost technology for the cohomological reduction of constrained Poisson algebras, introduced by Batalin, Fradkin and Vilkovisky [BF83, FF78, FV75], which extended the complex of BRST by adjoining odd generators, called ghosts and antighosts, thus reinventing the Koszul–Tate [Tat57] resolution of the ideal of constraints and producing a synergistic combination of both Chevalley– Eilenberg and resolution cohomology. Here it was that I saw the essential features of a strong homotopy Lie algebra (L∞ -algebra).

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J. Stasheff

5.1 Moment maps, momaps, and symplectic reduction The setting is one of Alan’s favorites [Wei02], that of a moment map, though generalized in an important way. Alan considers a phase space with a symmetry group consists of a manifold P equipped with a symplectic structure ω and a hamiltonian action of a Lie group G. By the latter, we mean a symplectic action of G on P together with an equivariant moment map J from P to the dual g∗ of the Lie algebra of G such that, for each v ∈ g, the one-parameter group of transformations of P generated by v is the flow of the hamiltonian vector field with hamilitonian x →< J (x), v >. The map J is called the momentum map (or, by many authors, moment map) of the hamiltonian action. If one is simply given a symplectic action of G on P , any map J satisfying the condition in italics above, even if it is not equivariant, is called a momentum map for the action. By contrast, Batalin–Fradkin–Vilkovisky consider constraints on the symplectic manifold P to be paramount. A Hamiltonian system with constraints means we have functions φα : P → R, 1 ≤ α ≤ r, the constraints. Solutions of the system are constrained to lie in a subspace V ⊂ P given as the zero set of a smooth momap φ : P → W = R r with components φα . In contrast to the more restrictive case in which W = R r has the structure of the dual of a Lie algebra g and φ is assumed to be equivariant with respect to the action of the corresponding Lie group on P , here we do not assume any Lie group G action. To emphaisze this, I refer to φ as a momap. (This also avoids the moment versus momentum controversy revealed to me last night.) The algebra C ∞ (V ) is given by C ∞ (P )/I , where I is the ideal generated by the φα . Dirac calls the constraints first class if I is closed under the Poisson bracket. In terms of the constraints, the condition is then γ

{φα , φβ } = fαβ φγ , γ

where we have structure functions fαβ on P , not structure constants. In other words, we have an analogue of a Lie algebroid with anchor map a : C ∞ (P ) → (T P ) given by the Hamiltonian vector field associated to a function. If we let W denote the vector space spanned by the φα , physicists speak of W as an open algebra since the bracket defined on W does not close in W . Compare this with Lie’s notion of function group [Lie90] as discussed by Alan [Wei02]. In this first class case, the Hamiltonian vector fields Xφα determined by the constraints are tangent to V (where V is smooth) and give a foliation F of V . Similarly, C ∞ (P )/I is an I -module with respect to the bracket. (In symplectic geometry, the corresponding variety is called coisotropic. The passage from P to V /F is known as symplectic reduction.) The true physics of the system is the induced system on the space of leaves V /F. If that space is a smooth manifold, C ∞ (V /F) is the true algebra of observables. When C ∞ (V /F) makes no sense, the Batalin–Fradkin–Vilkovisky construction provides a replacement, as described below (see [HT92] for a comprehensive treatment).

Poisson homotopy algebra

591

In this context, the classical BRST construction, at least as developed by Batalin– Fradkin–Vilkovisky in the case of regular constraints, is a homological model for C ∞ (V /F) or rather for the full de Rham complex (V , F) consisting of forms on vertical vector fields, those tangent to the leaves. The model is constructed as follows: First, consider the most common case of an equivariant moment map φ : P → W = g∗ with respect to a Lie group action of G on P , where g is the Lie algebra of G. Let A denote C ∞ (P ) considered as a Poisson algebra. Extend A as a graded commutative algebra to BFV = A ⊗ Eg∗ ⊗ Eg

(2)

and extend the Poisson bracket {·, ·} (still of degree 0) as determined by the fundamental pairing g∗ ⊗g → R. Note: Elements of g are called antighosts and have degree −1, while elements of g∗ are called ghosts and have degree 1. Now make BFV a dg Poisson algebra by defining dBFV = dK + δ ∗ , (3) where δ ∗ is the Chevalley–Eilenberg coboundary and dK is the Koszul differential on A ⊗ Eg regarded as a resolution of the ideal of constraints. In terms of a basis {eα } for g so that φα = eα ◦ φ, this means that dK is the graded derivation determined by dK (eα ) = φα . If we denote eα as Pα and define ηα in terms of a dual basis, then dBFV = {Q0 + Q1 , ·} for γ Q0 = ηα Pα and Q1 = 1/2ηα ηβ Cαβ Pγ , the formula that often appears in the physics literature. Because we have a strict Lie group action and, hence, structure constants, it is 2 = 0, but this is not the case for our momaps. The straightforward to verify dBFV definition of the algebra is no problem: BFV = A ⊗ EW ⊗ EW ∗

(4)

and dK + δ ∗ is defined as before but fails to square to 0, essentially because we now have structure functions. In the regular case, the brilliance of Batalin–Fradkin– Vilkovisky was to define dBFV by adding terms of higher order to dK + δ ∗ so that (dBFV )2 = 0. With hindsight, the existence of such terms of higher order was due to the fact that A ⊗ EW provided a resolution of the ideal of constraints, thus permitting the techniques of homological perturbation theory. However, the proof crucially involves keeping dBFV as an inner derivation {Q, ·} by adding terms of higher order to Q0 + Q1 . If we write Q = Q0 + Q∞ , then we see we are seeking a solution of the master equation (a.k.a. Maurer–Cartan) (see Section 6.3): {Q0 , Q∞ } + 1/2{Q∞ , Q∞ } = 0, or, equivalently, we seek to deform Q0 in the direction of Q1 (see Section 7). The point of doing this is as follows.

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Theorem 5.1. If the first class constraints generate a regular ideal, then the cohomology of BFV is isomorphic to the cohomology of (V , F) with respect to the leaf-wise exterior differential. In particular, H 0 (BFV) is isomorphic to H 0 ( (V /F)), the algebra of “observables’’ on the reduced phase space. In the more general nonregular case, the Koszul complex can be extended to the Koszul–Tate resolution by adding the polynomial algebra generated by “antighosts of antighosts’’ (given degree 2), etc. To preserve the crucial Poisson algebra structure, one also adds “ghosts of ghosts’’ (given degree −2), etc. In general, the quotient space is not a manifold, often not even Hausdorff, then H 0 (BFV) provides a suitable candidate for the algebra of observables on the “reduced phase space.’’ Since BFV is a free graded commutative algebra over A, assuming sufficient finiteness, the differential derivation dBFV is graded dual to a differential coderivation on a free graded cocommutative coalgebra over A and hence is equivalent to an L∞ -algebra. This is spelled out in considerable detail by Kjeseth [Kje01a, Kje01b], subsequent to some relevant observations by Huebschmann [Hue90] and myself.

6 Lagrangians with symmetries Lagrangian physics derives “equations of motion’’ from a variational principle of least action. Here an action refers to an integral S(φ) = L((j n φ)(x)) volM M

over some manifold M where φ is a (possibly vector valued) function on M or section of a bundle E over M. The action may have symmetries, i.e., variations in φ which do not change the value of S and hence are physically irrelevant in the sense that φ and its transformed value encode the same physical information. Emmy Noether had two major theorems regarding the variational calculus. The first, much better known and often referred to as Noether’s theorem, asserts a correspondence between symmetries and conserved quantities. Noether’s second variational theorem establishes a correspondence between symmetries, notably gauge symmetries, and differential algebraic relations among the Euler–Lagrange equations. It is this second theorem that has an important role in the Batalin–Vilkovisky construction for Lagrangians with symmetries. These symmetries create difficulties for quantization of such physical theories. The method of Batalin and Vilkovisky [BV84, BV83] was invented to handle these difficulties, but turns out to be of interest also in a classical context. The construction is quite parallel to that of Batalin–Fradkin–Vilkovisky in the constrained Hamiltonian case, but with one crucial difference: instead of a grading preserving bracket, they use an “antibracket’’ (independently due to Zinn-Justin [ZJ75, ZJ76]) which is of degree 1. Therefore, it is also known as an odd Poisson or Gerstenhaber bracket. In this Lagrangian setting, Batalin and Vilkovisky extend the BRST cohomological


593

approach by introducing antifields (independently and previously due to Zinn-Justin) dual to the original fields and antighosts which (with hindsight) correspond to the Noether relations and are dual to the ghosts which generate the BRST complex for the Lie algebra of symmetries. The original version of Noether in “Invariante Variationsprobleme’’ [Noe18] was written in terms of an infinite continuous group, G∞ρ , “understood to be a group whose most general transformations depend on ρ essential arbitrary functions and their derivatives.’’ Noether’s Theorem II refers to an integral I (= S in our notation) and reads as follows: If the integral I is invariant with respect to G∞ρ in which the arbitrary functions occur up to the σ th derivatives, there subsist ρ identity relationships between the Lagrange expressions and their derivatives up to the σ th order. . . . The converse holds. Later in that paper these relations are called dependencies. The relevance of Noether’s theorem is not emphasized in most of the literature using the BV approach. As with BFV, part of the differential of the Batalin– Vilkovisky complex BV is that of the Koszul–Tate resolution, in this case of the differential ideal generated by the Euler–Lagrange equations. The antifields generate the Koszul complex, which is not a resolution; the antighosts provide the next level of generators, as described by Tate [Tat57], corresponding to the relations among the Euler–Lagrange equations. It is the full acyclicity of the Koszul– Tate resolution that permits the application of homological perturbation theory [Gug82, GL89, GLS90, GS86, Hue84, HK91] and thus guarantees the existence of the terms of higher order in the full differential dBV . As in the concluding remark in Section 5, the graded dual to dBV is equivalent to an L∞ -algebra. We comment on this further in Section 6.2. Rather than carrying out this analysis in the abstract, we mention two particularly striking realizations of this structure: the Poisson sigma models of Cattaneo and Felder [CF99] and our analysis with Fulp and Lada [FLS02a, FLS02b] of Lagrangians with field dependent symmetries as in the case of higher spin particles. 6.1 The Poisson sigma model The fields of the Cattaneo–Felder σ -model are ordered pairs (X, η) such that X is a mapping from a two-dimensional manifold into a Poisson manifold M and η is a section of the bundle Hom(T , X∗ T ∗ M) −→ . These fields are subject to boundary conditions, namely they should satisfy the conditions X(u) = 0 and η(u)(v) = 0 for arbitrary u in the boundary of and for v tangent to the boundary of at u. Observe that for each u ∈ , we can regard η(u) as a linear mapping ∗ M. In local coordinates {uµ } on and {x i } on M, we write from Tu into TX(u) ∂ dX = (dXj ) ∂x j and η( ∂u∂ µ ) = ηi,µ dx i . The Poisson structure is given by a Poisson tensor α, which is a skew-symmetric tensor on M: ∂ ∂ α = α ij ∧ , (5) ∂x i ∂x j

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which satisfies a Jacobi condition: α il ∂l α j k + α j l ∂l α ki + α kl ∂l α ij = 0. The action S of the model is defined in such local coordinates by 1 S(X, η) = (ηi ∧ dX i ) + (α ij ◦ X)(ηi ∧ ηj ). 2

(6)

(7)

According to the variational principle, we obtain extrema of S as those fields (X, η) which satisfy the Euler–Lagrange equations 1 EXi := dηi + ∂i α j k (ηj ∧ ηk ) = 0 2

(8)

Eηi := −dXi − α ij ηj = 0.

(9)

and The gauge symmetries of the action are parameterized by all sections β of the bundle X∗ T ∗ M −→ which vanish on the boundary of . For each such β, define δβ acting on the fields by (δβ X)i = (α ◦ X)(dx i , β), (δβ η)(W ◦ X) = −(dβ)(W ◦ X) − ((LW α) ◦ X)(η, β),

(10) (11)

where W is a vector field on M, and LW α is the Lie derivative of α with respect to W . In terms of components of the fields, we write 1 EXi = (∂µ ηi,ν + ∂i α j k ηj,µ ηk,ν ) µν 2

(12)

Eηi,ν = −(∂µ X i + α ij ηj,µ ) µν .

(13)

and

It follows from Noether’s theorem that α ik EXi + ∂µ Eηk,µ − ∂i α j k ηj,µ Eηi,µ = 0

(14)

are the Noether identities corresponding to the gauge symmetry δβ defined above. Applied to this Poisson sigma model, the Batalin–Vilkovisky graded algebra BV is a graded commutative algebra over LocE (the algebra of local functions on E) with generators Xi+ and η+i , called “antifields,’’ γi , called “ghosts,’’ and γ +i , called “antighosts.’’ (If only the ghosts were added as generators, this would be just a BRST algebra.) These generators are bigraded. The graded commutativity is with respect to the sum (which we call the total degree) of the ghost degree and the form degree. The pairing between symmetries and identities is now expressed as the pairing between ghosts and antighosts, which plays a crucial role in the Batalin–Vilkovisky antibracket ( , ).


595

Now the initial differential on BV can be expressed as (S 0 + S 1 ), where S 0 is our original action and S 1 is 1 Xi+ α ij (X)γj − η+i ∧ (dγi + ∂i α kl (X)ηk γl ) − γ +i ∂i α j k (X)γj γk . (15) 2 Corresponding to the fact that (dKT + δ)2 = 0, as in BFV, we have (S 0 + S 1 , S 0 + S 1 ) = 0. Batalin and Vilkovisky show that, in much more general situations, one can add terms S i of ghost degree i > 1 to achieve a total SBV such that (SBV , SBV ) = 0. The reason for this is that the dKT homology vanishes in appropriate degrees, so the methods of homological perturbation theory apply again. In the Cattaneo–Felder model, only one more term is needed: 1 S2 = − η+i ∧ η+j ∂i ∂j α kl (X)γk γl . (16) 4 Thus the total Batalin–Vilkovisky generator SBV is 1 ηi ∧ dX i + α ij (X)ηi ∧ ηj 2 1 + Xi+ α ij (X)γj − η+i ∧ (dγi + ∂i α kl (X)ηk γl ) − γ +i ∂i α j k (X)γj γk 2 1 +i +j kl − η ∧ η ∂i ∂j α (X)γk γl . (17) 4 6.2 Field dependent gauge symmetries Field dependent gauge symmetries appear in several field theories, most notably in a class due to Ikeda [Ike94] and Schaller and Strobl [SS94], including the Poisson sigma model of Cattaneo and Felder [CF99] above. A significant generalization occurs in the Berends, Burgers, and van Dam [Bur85, BBvD86, BBvD85] approach to “particles of spin ≥ 2.’’ The physics of “particles of spin ≤ 2’’ leads to representations of a Lie algebra + of gauge parameters on a vector space of fields. By a field dependent action of + on , Berends, Burgers, and van Dam mean a polynomial (or power series) map δ(ξ )(φ) = i≥0 Ti (ξ, φ), where Ti is linear in ξ and polynomial of homogeneous degree i in φ. Berends, Burgers, and van Dam consider arbitrary field theories, subject only to the requirement that the commutator of two gauge symmetries be another gauge symmetry whose gauge parameter is possibly field dependent. Thus they do not require an a priori given Lie structure to induce the algebraic structure of the gauge symmetry “algebra.’’

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Let denote the vector space of fields and + the vector space of gauge parameters. Let ∗ denote the free graded cocommutative coalgebra cogenerated by . Although the space + of gauge parameters has no natural Lie structure, the space of linear maps from ∗ into + is a Lie algebra under certain mild assumptions along with a hypothesis which we refer to as the BBvD hypothesis. Under these assumptions, the gauge algebra gives rise to an L∞ -algebra on a differential graded vector space V with + in degree 0, in degree 1 and 0 in all other degrees. The vector space Coder(∗ ) of coderivations on ∗ is a Lie algebra with bracket given by the commutator with respect to composition. The vector space Hom(∗ , ) is isomorphic to Coder(∗ ) and hence inherits a Lie algebra structure; the bracket on Hom(∗ , ) is known as the Gerstenhaber bracket [Ger63, Sta93]. Suppose that we are given a linear map δ : + → Hom(∗ , ), a “field dependent action’’ of + on . By a field dependent action of + on , Berends, Burgers, and van Dam [Bur85, BBvD84, BBvD85] mean a polynomial (or power series) map δ(ξ )(φ) = i=0 Ti (ξ, φ) where Ti is linear in ξ and polynomial of homogeneous degree i in φ. We adopt the corresponding polarized and adjoint point of view and write δ(ξ ) = i=0 Ti (ξ ) where Ti is zero except on i . We extend δ to a map δˆ : Hom(∗ , +) → Hom(∗ , ) by

ˆ δ(π) = ev ◦ (δ ◦ π ⊗ 1) ◦

,

where ev is the evaluation map. Consider the possibility of inducing a Lie-type bracket ˆ Under certain conditions, e.g., δ is injective, on Hom(∗ , +) via the mapping δ. such a bracket may then be used to obtain a bracket on the parameter space + by restricting the bracket on Hom(∗ , +), where we think of + as being contained in the space Hom(∗ , +) by identifying ξ ∈ + with the map (also denoted ξ ) in Hom(∗ , +), which is 0 except on the scalars, where ξ(1) = ξ . In order to assure the Jacobi property of the bracket on Hom(∗ , +), we introduce a correction term. We accomplish this, following Berends, Burgers, and van Dam, by assuming there is a map C : + ∧ + → Hom(∗ , +) such that

[δ(ξ ), δ(η)] = δC(ξ, η) ∈ Hom(∗ , )

for all ξ, η ∈ +. We refer to this as the BBvD hypothesis. We then extend C to a mapping Cˆ : Hom(∗ , +) ∧ Hom(∗ , +) → Hom(∗ , +) by

ˆ 1 , π2 ) = C ◦ ((π1 ⊗ π2 ) ⊗ 1) ◦ ( C(π

⊗ 1) ◦

,

where we have identified C with its adjoint mapping, the mapping from +⊗+⊗∗ into + defined by (ξ, η, φ1 ∧ · · · ∧ φn ) −→ C(ξ, η)(φ1 ∧ · · · ∧ φn ).


597

Next, we redefine the bracket on Hom(∗ , +) by including the correction term ˆ 1 , π2 ). [π1 , π2 ] = π1 δ(π2 ) − π2 δ(π1 ) + C(π

(18)

ˆ 1 , π2 ] = [δ(π1 ), δ(π2 )]. Theorem 6.1. The mapping δˆ preserves brackets, that is, δ[π ∗ ∗ Moreover, if δ : Hom( , +) → Hom( , ) is injective, then [π1 , π2 ] satisfies the Jacobi identity. This suggests that the parameter space should be enlarged to include all of Hom(∗ , +), but this is apparently unacceptable to physicists since the number of independent parameters is linked to the number of independent Noether identities. However, the polynomial equations of physical relevance define an L∞ -structure on an appropriate graded vector space. We restrict our attention to the constant maps in Hom(∗ , +) and show that the algebraic structure of Hom(∗ , +) induces an L∞ -structure on + ⊕ . We assume the hypothesis and that δˆ is injective so Theorem 6.1 holds. Define a differential graded vector space V with + in degree 0, in degree 1, and 0 in all other degrees. Take ∂ : + → , given by ∂(ξ ) = δ(ξ )(1) ∈ , as the only nontrivial differential. Define D : ∗ (sV ) → sV by D(ξ ) = ∂(ξ ), D(ξ ∧ φ1 ∧ · · · ∧ φn ) = δ(ξ )(φ1 ∧ · · · ∧ φn )

for n ≥ 1,

D(ξ1 ∧ ξ2 ∧ φ1 ∧ · · · ∧ φn ) = C(ξ1 , ξ2 )(φ1 ∧ · · · ∧ φn ), and D = 0 on elements of ∗ (sV ) with more than two entries from + or with no entry from +. Notice this is essentially not of the same form as that of Roytenberg and Weinstein in Section 4.2, although both have just two components. The crucial difference is in the grading: 0, 1 here versus −1, 0 for them. Theorem 6.2 ([FLS02a]). D : ∗ (sV ) → sV as defined above gives V the structure of an L∞ -algebra. 6.3 The master equation and homological perturbation theory The name “master equation’’ derives from the physics literature, especially of the Batalin–Vilkovisky approach considered above, but equations of this form are well known in mathematics, though under various names: • • •

the defining equation for a twisting cochain, the integrability equation of deformation theory, the Maurer–Cartan equation;

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the latter is perhaps the most famous. The equation makes sense as applied to elements of a dg algebra, associative or Lie or Gerstenhaber, etc., and has generalizations to higher homtopy versions. In [HS02], Huebschmann and I give an extensive comparison of these various interpretations. We show how to construct solutions using the tools of homological perturbation theory, working in characteristic zero. In particular, we endow the homology H (g) of a strict dg Lie algebra g with the structure of an L∞ -algebra such that g and H (g) are equivalent as L∞ -algebras, i.e., via L∞ maps (see Section 7). The much older analogous result for A∞ -algebras is due to Kadeishvili [HK91]. Note that H (g) is a strict dg Lie algebra with d = 0, but the higher-order operations li are often nontrivial. If g is equivalent as L∞ -algebra to H (g) with all li = 0 for i ≥ 3, then g is called formal.

7 L∞ -maps, deformation quantization, string field theory (SFT), and more Definition 7.1. An L∞ -map f : h → g of L∞ -algebras (or dgLie algebras) is a dg coalgebra map c (sh) → c (sg). The Cattaneo and Felder Poisson sigma model was developed to provide an alternative, “path integral,’’ proof of Kontsevich’s theroem that any Poisson manifold can be deformation quantized. In both proofs, the key issue is the formality of a certain dgLie algebra g. The L∞ -equivalence of this g and H (g) implies that all the obstructions to deformation quantization vanish. For this important application, was a disk so the maps → M could be considered as world sheets as in SFT. Because BBvD give an explicit expansion Ti , Ci , the corresponding multi-brackets li are visible or at least easy to extract. In contrast, in the Cattaneo and Felder Poisson sigma model, they are hidden in the single function α and its derivatives. The relevance of A∞ - and L∞ -structure to (respectively) OSFT and CSFT has a particularly “physical’’ interpretation. The higher order operations describe multiple string interactions, not obtained from three-string interactions (multiplication, respectively, bracketing of two strings) or the equivalent correlation functions [Zwi93]. Here too there is contact with Alan and his student Tang in their recent paper [TW04]. A combined open-closed string field theory [Zwi98] leads to an intricate combination of an L∞ -algebra acting by strong homotopy derivations of an A∞ -algebra [HK91].

8 Homological Legendre transform In their concluding remarks in [RW98], Dmitry and Alan muse: L∞ -algebras occur in physics in the framework of the Batalin–Vilkovisky procedure for quantizing gauge theories. On the other hand, the Courant bracket seems to provide a geometric framework for constrained Hamiltonian


599

systems. It is known [HT92] that gauge Lagrangians lead to constrained theories in the Hamiltonian formalism. This suggests that homotopy Lie algebras arising in the Batalin–Vilkovisky formalism and those in the Courant formalism might be somehow related. In response to my paper for the Alanfestschrift, Dmitry pointed out to me the paper of Grigoriev and Damgaard which establishes an analogue of the Legendre transform in terms of the BFV and BV constructions. Here at Alanfest, we have investigated their transforms in further detail. This bears further investigation, but for now let me mention only that in either direction, Hamiltonian to Lagrangian of vice versa, the essential idea is the “oddification’’ of all the fields, ghosts, etc., then substituting these into the respective formulas for the Hamiltonian, the Lagrangian, etc., and keeping only the parts of the appropriate total degree. Dmitry can interpret this further by looking at the algebra as that of a graded path space.

9 Coda There are still other examples of A∞ - and L∞ -structures with potential physical relevance, for example, the notion of A∞ -category. A∞ -categories have been used by Fukaya [Fuk95] for remarkable applications to Morse theory and Floer homology. More recently, they play a role in string and D-brane theory and homological mirror symmetry. But that takes us further afield from today’s topic: the L∞ -structures directly involved in some of Alan’s work and closely related to his foundational work on symplectic reduction. There are further relations to be discovered, as he has indicated. Leaving that for the future, let me conclude with best wishes for the continuation of a long happy and inspiring career to Alan on his 60th birthday.

References [BBvD84] F. A. Berends, G. J. H. Burgers, and H. van Dam, On spin three selfinteractions, Z. Phys. C, 24 (1984), 247–254. [BBvD85] F. A. Berends, G. J. H. Burgers, and H. van Dam, On the theoretical problems in constructing intereactions involving higher spin massless particles, Nuclear Phys. B, 260 (1985), 295–322. [BBvD86] F. A. Berends, G. J. H. Burgers, and H. van Dam, Explicit construction of conserved currents for massless fields of arbitrary spin, Nuclear Phys. B, 271 (1986), 429–441. [BF83] I. A. Batalin and E. S. Fradkin, A generalized canonical formalism and quantization of reducible gauge theories, Phys. Lett., 122B (1983), 157–164. [BRS75] C. Becchi, A. Rouet, and R. Stora, Renormalization of the abelian Higgs-Kibble model, Comm. Math. Phys. 42 (1975), 127–162. [Bur85] G. J. H. Burgers, On the Construction of Field Theories for Higher Spin Massless Particles, Ph.D. thesis, Rijksuniversiteit te Leiden, Leiden, the Netherlands, 1985. [BV83] I. A. Batalin and G. S. Vilkovisky, Quantization of gauge theories with linearly dependent generators, Phys. Rev. D, 28 (1983), 2567–2582.

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I. A. Batalin and G. S. Vilkovisky, Closure of the gauge algebra, generalized Lie equations and Feyneman rules, Nuclear Phys. B, 234 (1984), 106–124. [BC03] J. C. Baez andA. S. Crans, Higher-dimensional algebra VI: Lie 2-algebras, preprint, 2003; math.QA/0307263. [CE48] C. Chevalley and S. Eilenberg, Cohomology theory of Lie groups and Lie algebras, Trans. Amer. Math. Soc., 63 (1948), 85–124. [CF99] A. Cattaneo and G. Felder, A path integral approach to the Kontsevich quantization formula, Comm. Math. Phys., 212-3 (2000), 591–611 [Dai02] M. Daily, L-infinity structures on spaces with 3 one-dimensional components, preprint, 2002; math.QA/0212030. [FF78] E. S. Fradkin and T. E. Fradkina, Quantization of relativistic systems with boson and fermion first and second class constraints, Phys. Lett., 72B (1978), 343–348. [FLS02a] R. Fulp, T. Lada, and J. Stasheff, Noether’s variational theorem II and the BV formalism, Suppl. Rend. Circ. Mat. Palermo Ser. II, 71 (2002), 115–126. [FLS02b] R. Fulp, T. Lada, and J. Stasheff, Sh-Lie algebras induced by gauge transformations, Comm. Math. Phys., 231 (2002), 25–43. [FP67] L. D. Fade’ev and V. N. Popov, Feynman diagrams for the Yang-Mills field, Phys. Lett., 25B (1967), 29–30. [FP03] A. Fialowski and M. Penkava, Versal deformations of three dimensional lie algebras as L-infinity algebras, preprint, 2003; math.RT/0303346. [Fuk95] K. Fukaya, Floer homology, A∞ -categories and topological field theory, in J. Andersen, J. Dupont, H. Pertersen, and A. Swan, eds., Geometry and Physics, Lecture Notes in Pure and Applied Mathematics, Vol. 184, Marcel Dekker, New York, 1995, 9–32 (notes by P. Seidel). [FV75] E. S. Fradkin and G. S. Vilkovisky, Quantization of relativistic systems with constraints, Phys. Lett., 55B (1975), 224–226. [Ger63] M. Gerstenhaber, The cohomology structure of an associative ring, Ann. Math., 78 (1963), 267–288. [GL89] V. K. A. M. Gugenheim and L. Lambe, Applications of perturbation theory to differential homological algebra I, Illinois J. Math., 33 (1989), 556–582. [GLS90] V. K. A. M. Gugenheim, L. Lambe, and J. Stasheff, Algebraic aspects of Chen’s twisting cochain, Illinois J. Math., 34 (1990), 485–502. [GS86] V. K. A. M. Gugenheim and J. D. Stasheff, On perturbations and A∞ -structures, Bull. Soc. Math. Belgium, 38 (1986), 237. [Gug82] V. K. A. M. Gugenheim, On a perturbation theory for the homology of a loop space, J. Pure Appl. Algebra, 25 (1982), 197–207. [HK91] J. Huebschmann and T. Kadeishvili, Small models for chain algebras, Math. Z., 207 (1991), 245–280. [HS02] J. Huebschmann and J. Stasheff, Formal solution of the master equation via HPT and deformation theory, Forum Math., 14 (2002), 847–868. [HT92] M. Henneaux and C. Teitelboim, Quantization of Gauge Systems, Princeton University Press, Princeton, NJ, 1992. [Hue84] J. Huebschmann, Perturbation Theory and Small Models for the Chains of Certain Induced Fibre Spaces, Habilitationsschrift, 1984. [Hue90] J. Huebschmann, Poisson cohomology and quantization, J. Reine Angew. Math., 408 (1990), 57–113. [Ike94] N. Ikeda, Two-dimensional gravity and nonlinear gauge theory, Ann. Phys., 235 (1994), 435–464. [Kaj03] H. Kajiura, Noncommutative Homotpy Algebras Associated with Open Strings, Dissertation, University of Tokyo, Tokyo, 2003.

Poisson homotopy algebra [Kje01a] [Kje01b] [KS03]

[Lie90] [MSS02]

[Nas98] [Noe18]

[RW98] [SS94] [Sta93]

[Sto77] [Tat57] [TW04] [Tyu75] [Wei02] [ZJ75]

[ZJ76]

[Zwi93] [Zwi98]

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L. Kjeseth, A homotopy Lie-Rinehart resolution and classical BRST cohomology, Homology Homotopy Appl., 3-1 (2001), 165–192 (electronic). L. Kjeseth, Homotopy Rinehart cohomology of homotopy Lie-Rinehart pairs, Homology Homotopy Appl., 3-1 (2001), 139–163 (electronic). Y. Kosmann-Schwarzbach, Quasi, twisted, and all that… in Poisson geometry and Lie algebroid theory, in J. E. Marsden and T. S. Ratiu, eds., The Breadth of Symplectic and Poisson Geometry: Festschrift in Honor of Alan Weinstein (this volume), Progress in Mathematics, Vol. 232, Birkhäuser, Boston, 2005, 363–390. S. Lie, Theorie der Tranformationensgruppen, Teubner, Leipzig, 1890. M. Markl, S. Shnider, and J. Stasheff, Operads in Algebra, Topology and Physics, Mathematical Surveys and Monographs, Vol. 96, American Mathematical Society, Providence, RI, 2002. C. Nash, Topology and physics: A historical essay, in I. M. James, ed., A History of Topology, Elsevier–North Holland, Amsterdam, 1998, 359–415. E. Noether, Invariante variationsprobleme, Nachr. König. Gesell. Wissen. Göttingen Math.-Phys. Kl., (1918), 235–257 (in German); Transport Theory Stat. Phys., 1 (1971), 186–207 (in English). D. Roytenberg and A. Weinstein, Courant algebroids and strongly homotopy Lie algebras, Lett. Math. Phys., 46-1 (1998), 81–93. P. Schaller and T. Strobl, Poisson structure induced (topological) field theories, Mod. Phys. Lett. A, 9 (1994), 3129–3136. J. D. Stasheff, The intrinsic bracket on the deformation complex of an associative algebra, J. Pure Appl. Algebra, 89 (1993) (festschrift in honor of Alex Heller), 231–235. R. Stora, Continuum gauge theories, in M. Levy and P. Mitter, eds., New Developments in Quantum Field Theory, Plenum, New York, 1977, 201–224. J. Tate, Homology of Noetherian rings and local rings, Illinois J. Math., 1 (1957), 14–27. X. Tang and A. Weinstein, Quantization and morita equivalence for constant dirac structures on tori, Ann. Inst. Fourier, 54 (2004), to appear; math.QA/0305413. I. V. Tyutin, Gauge invariance in field theory and statistical physics in operator formulation, technical report, Lebedev Physics Institute, Moscow, 1975 (in Russian). A. Weinstein, The Geometry of Momentum, 2002, math.SG/0208108. J. Zinn-Justin, Renormalization of gauge theories, in H. Rollnick and K. Dietz, eds., Trends in Elementary Particle Theory, Lecture Notes in Physics, Vol. 37, Springer-Verlag, 1975, 2–39. J. Zinn-Justin and R. Balian, eds., Méthodes en théorie des champs = Methods in Field Theory, North-Holland, Amsterdam, 1976 (École d’Été de Physique Théorique, Session XXVIII, tenue à Les Houches, 28 Juillet–6 Septembre, 1975). B. Zwiebach, Closed string field theory: Quantum action and the BatalinVilkovisky master equation, Nuclear Phys. B, 390 (1993), 33–152. B. Zwiebach, Oriented open-closed string theory revisited, Ann. Phys., 267 (1998), 193–248.

Dirac submanifolds of Jacobi manifolds Izu Vaisman Department of Mathematics University of Haifa 31905 Haifa Israel [email protected] Dedicated to Alan Weinstein on the occasion of his sixtieth birthday. Abstract. The notion of a Dirac submanifold of a Poisson manifold studied by Xu is interpreted in terms of a general notion of tensor fields soldered to a normalized submanifold. This interpretation is used to define the notion of a Dirac submanifold of a Nambu–Poisson and Jacobi manifold. Several properties and examples are discussed.

1 Normalized submanifolds In this section we make some general considerations on submanifolds of a differentiable1 manifold. These considerations were inspired by the theory of Dirac submanifolds of a Poisson manifold developed in [10]. The notion of a normalized submanifold was used in affine and projective differential geometry half a century ago. Definition 1.1. Let N n be a submanifold of M m (indices denote dimensions) and ι : N ⊆ M the corresponding embedding. A normalization of N by a normal bundle νN is a splitting T M|N = T N ⊕ νN (1) (T denotes tangent bundles). A submanifold endowed with a normalization is called a normalized submanifold. Then if X ∈ T M ( denotes spaces of global cross-sections) is a vector field on M such that X|N ∈ T N , respectively X|N ∈ νN , X is said to be tangent, respectively, normal, to N. Let (N n , νN) be a normalized submanifold of M m . Let σ : W → N be a tubular neighborhood of N such that ∀x ∈ N , Tx (Wx ) = νx N (Wx is the fiber of W and νx N is the fiber of νN at x). Then W is said to be a compatible tubular neighborhood of N ; obviously, such neighborhoods exist. Furthermore, each 1 In this paper, everything is of class C ∞ and all submanifolds are embedded.

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point x ∈ N has a σ -trivializing neighborhood U endowed with coordinates (x a ) (a, b, c, · · · = 1, . . . , m − n) on the fibers of σ and such that x a |N ∩U = 0, and coordinates (y u ) (u, v, w, · · · = m − n + 1, . . . , m) on N ∩ U . We will say that (x a , y u ) are adapted local coordinates. With respect to adapted coordinates, N has the local equations x a = 0, and ∂ ∂ T N|U ∩N = span , νN | . (2) = span U ∩N ∂y u x a =0 ∂x a x a =0 Accordingly, the transition functions between two systems of adapted local coordinates must be of the form x˜ a = x˜ a (x b , y v ),

y˜ u = y˜ u (y v ),

(3)

and satisfy the conditions ∂ x˜ a = 0, ∂y v x b =0

∂ y˜ u ≡ 0. ∂x b

(4)

The splitting (1) induces a similar relation for the dual bundles T ∗ M|N = T ∗ N ⊕ ν ∗ N,

(5)

and locally, with respect to adapted coordinates, one has T ∗ N = ann(νN ) = span{dy u |x a =0 }, ν ∗ N = ann(T N ) = span{dx a |x a =0 }

(6)

(ann denotes annihilator spaces). Two normal bundles νN and ν˜ N of the same submanifold N are connected as follows. Let pν , pT be the projections defined by the splitting (1) and pν˜ , p˜ T the similar projections of the second normalization. The mapping (v ∈ νN ) → pν˜ v is an isomorphism ϕ : νN → ν˜ N , and with respect to adapted coordinates, we have ∂ c ν˜ N = span ϕ | = X (7) a x =0 , ∂x a x c =0 where2 Xa =

∂ ∂ − θau u ∂x a ∂y

(8)

are vector fields on U , and (θau |x c =0 ) is the local matrix of the homomorphism ψ : νN → T N defined by ψ(v) = p˜ T (v) (v ∈ νN ). Notice that ϕ + ψ is the inclusion of νN in T M|N , and ν˜ N is uniquely determined by any of the mappings ϕ, ψ. Some geometric objects of M may have a strong relationship with the normalized submanifold (N, νN ). 2 In this paper, we use the Einstein summation convention.

Dirac submanifolds of Jacobi manifolds

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Definition 1.2. A differential k-form κ ∈ k (M) ( denotes spaces of differential forms) is soldered to N if ι∗ [LX κ] = 0 for any vector field X ∈ T M normal to N . Since ∀f ∈ C ∞ (M) and any vector fields X, Y1 , . . . , Yk , one has (Lf X κ)(Y1 , . . . , Yk ) = f (LX κ)(Y1 , . . . , Yk ) −

k

(9)

(−1)j (Yj f )[i(X)κ](Y1 , . . . , Yj −1 , Yj +1 , . . . , Yk ),

j =1

it follows that κ is soldered iff for any vector field X ∈ T M normal to N , one has ι∗ [i(X)κ] = 0,

ι∗ [LX κ] = 0,

(10)

ι∗ [i(X)κ] = 0,

ι∗ [i(X)dκ] = 0.

(11)

or, equivalently,

With respect to adapted local coordinates, κ has the expression κ=

s+t=k

1 κa ...a u ...u dx a1 ∧ · · · ∧ dx as ∧ dy u1 ∧ · · · ∧ dy ut , s!t! 1 s 1 t

and κ is soldered to N iff κau1 ...uk−1 |x b =0 = 0,

∂κu1 ...uk = 0. ∂x a x b =0

(12)

(13)

In particular, the space of soldered functions is C ∞ (M, N, νN) = {f ∈ C ∞ (M) /(∂f/∂x a )x a =0 = 0}.

(14)

We will denote by k (M, N, νN) the space of soldered k-forms (for k = 0 we have the space (14)). Obviously, the soldering conditions (11) are compatible with the exterior product and the exterior differential. Therefore, we get a cohomology k (M, N, νN), which will be called the soldered de Rham cohomolalgebra ⊕k HsdeR ogy algebra, defined by the cochain spaces k (M, N, νN) and the operator d. The inclusion in the usual de Rham complex induces homomorphisms k k ιk : HsdeR (M, N, νN) −→ HdeR (M).

(15)

k (W, N, νN), where W is a compatible tubular neighIn principle, the spaces HsdeR borhood, should provide interesting information about the normalized submanifold (N, νN).

Definition 1.3. A k-vector field Q ∈ V k (M) (V denotes spaces of multivector fields) is soldered to the normalized submanifold (N, νN ) if

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(i) for any (k − 1)-form λ ∈ ∧k−1 [ann(νN )], the vector field defined along N by i(λ)Q|N is tangent to N ; (ii) for any vector field X on M normal to N , (LX Q)|ann(νN ) = 0. We will denote by V k (M, N, νN) the space of soldered k-vector fields. Using adapted local coordinates, we see that V 0 (M, N, νN) is, again, (14), and for k = 1 one has ∂ηu 1 1 u ∂ V (M, N, νN) = Y ∈ V (M) / Y |N = η , =0 . (16) ∂y u N ∂x a x c =0 Generally, we have an expression of the form Q=

s+t=k

1 a1 ...as u1 ...ut ∂ ∂ ∂ ∂ Q ∧ ··· ∧ a ∧ u ∧ ··· ∧ u , s!t! ∂x a1 ∂x s ∂y 1 ∂y t

and Q ∈ V k (M, N, νN) iff Qau1 ...uk−1 |x c =0 = 0,

∂Qu1 ...uk−1 c = 0. ∂x a x =0

(17)

(18)

The spaces of soldered forms and multivector fields are components of important algebraic structures; namely, we have the following. Proposition 1.1. 1. The space V 1 (M, N, νN) is a Herz–Reinhart Lie algebra over (R, C ∞ (M, N, νN )). 2. The complex of N-soldered differential forms is a complex over the Lie algebra V 1 (M, N, νN). 3. The triple (⊕k V k (M, N, νN), ∧, [ , ]), where [ , ] is the Schouten–Nijenhuis bracket is a Gerstenhaber algebra. Proof. For the definition of the algebraic structures above, see, for instance, [2] and [3]. The use of adapted local coordinates shows that if f ∈ C ∞ (M, N, νN) and Y, Z ∈ V 1 (M, N, νN), then f Y and [Y, Z] belong to V 1 (M, N, νN), which proves 1. Furthermore, for the same Y and any κ ∈ k (M, N, νN), i(Y )κ ∈ k−1 (M, N, νN), and we get 2. Finally, the exterior product of soldered multivector fields is obviously soldered, and in order to get 3, it remains to prove that the Schouten– Nijenhuis bracket3 of P ∈ V p (M, N, νN) and Q ∈ V q (M, N, νN) belongs to V p+q−1 (M, N, νN). To see that soldering condition (i) is satisfied, we look at the known formula (e.g., [8]) i([P , Q])ω = (−1)(p+1)(q+1) i(P )d[i(Q)ω] − i(Q)d[i(P )ω] + (−1)p i(P ∧ Q)dω,

(19)

3 We take this bracket with the sign convention of the axioms of graded Lie algebras, e.g., [8,

Proposition 4.21].


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where ω is an arbitrary (p + q − 1)-form on M, and use this formula for ω = dx a ∧ dy u1 ∧ · · · ∧ dy up+q−2 . Then soldering condition (ii) follows by using (19) to evaluate the terms of the equality LX [P , Q] = [LX P , Q] + [P , LX Q], where X is normal to N , on dy u1 ∧ · · · ∧ dy up+q−1 .

The following proposition extends a result proven for Poisson bivector fields in [10]. Proposition 1.2. If the involutive diffeomorphism ϕ : M → M (ϕ 2 = Id) preserves a k-form κ, respectively, a k-vector field Q, then κ, respectively, Q, is soldered to the fixed point locus N of ϕ. Proof. It is well known that N is a submanifold of M, the tangent bundle T N consists of the (+1)-eigenspaces of ϕ∗ along N , and N has a normalization with the normal bundle νN defined by the (−1)-eigenspaces of ϕ∗ along N [10]. This also implies that ann(νN) = T ∗ N consists of the (+1)-eigenspaces, and ann(T N ) = ν ∗ N consists of the (−1)-eigenspaces, of ϕ ∗ along N . If ϕ ∗ κ = κ, if X is a normal vector field of N on M and Y1 , . . . , Yk−1 are tangent to N , then κ(X, Y1 , . . . , Yk−1 )|N = (ϕ ∗ κ)(X, Y1 , . . . , Yk−1 )|N = −κ((X, Y1 , . . . , Yk−1 )|N ; hence ι∗ [i(X)κ] = 0. The same holds for dκ; therefore, κ is soldered to N . The proof for a k-vector field Q is similar, and uses the fact that ϕ∗ (LX Q) = Lϕ∗ X (ϕ∗ Q) ◦ ϕ for any diffeomorphism ϕ : M → N .

The N-soldered differential forms and multivector fields have a nice interpretation by means of the geometry of the tangent bundle T M, and by looking at the normal bundle νN as a submanifold of the former. (See [10] for the case of a Poisson bivector field.) The tensor fields of the manifold M may be lifted to T M by various processes and, in particular, there exists a complete lift, which comes from the lift of the flow of a vector field [11]. In the case of differential forms and multivector fields, the complete lift has the coordinate expression 1 κi ...i d z˙ i1 ∧ dzi2 ∧ · · · ∧ dzik (k − 1)! 1 k 1 ∂κi1 ...ik i1 + z˙ j dz ∧ · · · ∧ dzik , k! ∂zj 1 ∂ ∂ ∂ Qi1 ...ik i ∧ i ∧ · · · ∧ i QC = 1 2 (k − 1)! ∂z ∂ z˙ ∂ z˙ k ...i i 1 ∂Q 1 k ∂ ∂ + z˙ j ∧ ··· ∧ i . j i 1 k! ∂z ∂ z˙ ∂ z˙ k κC =

(20)

(21)

In formulas (20) and (21) κ and Q are given by the expressions (12) and (17), respectively, while (zi ) = (x a , y u ) (i = 1, . . . , m), and (˙zi ) are the corresponding natural vector coordinates.

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Proposition 1.3. (i) The differential form κ is soldered to the normalized submanifold (N, νN ) of M iff ∀Z ∈ T (νN), the form i(Z)κ C belongs to the ideal generated by [ann(T (νN ))]. (ii) The k-vector field Q is soldered to (N, νN ) iff ∀α ∈ [ann(T (νN ))], i(α)QC belongs to the ideal generated by T (νN). Proof. On M, we use N-adapted local coordinates and on T M the corresponding natural vector coordinates as described above. Then the submanifold νN has the local equations x a = 0, y˙ u = 0, and the results are immediate consequences of formulas (20) and (21).

We remark that it is possible to define soldered symmetric tensor fields, similarly. The following proposition provides a nice example. Proposition 1.4. Let M be a Riemannian manifold with the metric tensor g. Then g is soldered to a submanifold N normalized by the normal bundle νN ⊥ T N iff N is a totally geodesic submanifold. Proof. If ∇ is the Levi-Civita connection of g, i.e., ∇g = 0 and ∇ has no torsion, one has (LX g)(Y, Z) = g(∇Y X, Z) + g(Y, ∇Z X). Then if X is normal and Y, Z are tangent to N, the restriction of the previous formula to N yields (LX g)(Y, Z) = 2g(b(Y, Z), X), (22) where b is the second fundamental form of the submanifold N . Thus the soldering condition of g is equivalent to b = 0.

The notion of soldering has other interesting extensions, too. First, for a multivector field Q ∈ V k (M), condition (ii) of Definition 1.3 is itself a geometric condition, since it is easy to check that if it holds for X normal to N , it also holds for f X ∀f ∈ C ∞ (M). If Q satisfies only this condition, we will call it quasi-soldered to (N, νN). In fact, this notion extends to any contravariant tensor field. The notion of a soldered differential form also extends to any covariant tensor field, but it implies algebraic conditions like the first condition in (10) as well. Then we may look at objects that only satisfy the algebraic condition of soldering (e.g., the first condition (10), condition (i) of Definition 1.3, etc.), and call them algebraically compatible with the normalized submanifold . If the algebraic condition holds, the Lie derivative in the normal directions yields an important object for the submanifold. For instance, a Riemannian metric is algebraically compatible with any submanifold N , if the normal bundle is the g-orthogonal bundle of T N, and formula (22) shows that (LX g)|T N is equivalent to the second fundamental form of the submanifold. Finally, we may add to the algebraic condition a condition that is weaker than soldering. For instance, a tensor field that is algebraically compatible with a normalized submanifold will be called weakly soldered if, along the submanifold, the


609

Lie derivative in the normal directions are proportional to the pullback of the tensor field to the submanifold. For instance, the Riemannian metric g is weakly soldered to a submanifold N with the g-normal bundle if, for some 1-form α, one has (LX g)|T N = α(X)g|T N , for any normal vector field X, and this happens iff N is a totally umbilical submanifold.

2 Dirac submanifolds of Poisson and Nambu–Poisson manifolds In this section, we recall the definition and characteristic properties of the Dirac submanifolds of a Poisson manifold studied by Xu [10], and give a few additional facts. In particular, we extend Xu’s definition to Nambu–Poisson manifolds. We refer to [8] for generalities of Poisson geometry and to [9] for the Nambu–Poisson geometry. A Dirac submanifold of a Poisson manifold inherits an induced Poisson structure, and the cotangent Lie algebroid of the latter may be seen as a Lie subalgebroid of the cotangent Lie algebroid of the original manifold. Definition 2.1. A submanifold N n of a Poisson manifold M m , with the Poisson bivector field $, is a Dirac submanifold if N has a normalization (1) with the following properties: (i) $ (ann(νN)) ⊆ T N ($ is the morphism T ∗ M → T M defined by $); if this condition holds, we will say that νN is algebraically $-compatible; (ii) ∀x ∈ N, there exists an open neighborhood U of x in M such that ∀f, g ∈ C ∞ (U ) which satisfy the conditions df |νN = 0, dg|νN = 0 one has d{f, g}|νN = 0. ({f, g} is the Poisson bracket defined by $.) Proposition 2.1 ([10]). With the notation of Definition 2.1, the submanifold N is a Dirac submanifold iff there exists a normalization (1) such that the Poisson bivector field $ is soldered to (N, νN ). Proof. $ is soldered to (N, νN ) iff with the notation and the adapted coordinates as defined in Section 1, one has $=

∂ ∂ 1 ∂ ∂ ∂ 1 ab ∂ $ ∧ b + $au a ∧ u + $uv u ∧ v , a 2 ∂x ∂x ∂x ∂y 2 ∂y ∂y

(23)

where $au |x c =0 = 0, ∂$uv = 0. ∂x a c

(24) (25)

x =0

On the other hand, if $ is given by (23), condition (i) of Definition 2.1 is equivalent to $ (dy u ) ∈ span{∂/∂y v } along N , which means (24), and condition ii) is equivalent

to the fact that d{y u , y v }|x c =0 = 0, which is (25). Furthermore, from the definition of soldered multivector fields, we also get the following.

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Proposition 2.2 ([10]). The submanifold N of (M, $) is a Dirac submanifold iff N has a $-compatible normal bundle νN such that for any normal to N vector field X of M, one has (LX $)|ann(νN ) = 0. (26) Corollary 2.1. Let {Xα } be a family of Poisson infinitesimal automorphisms of (M, $). Then any submanifold N such that span{Xα |N } is a $-compatible normal bundle of N is a Dirac submanifold. Proof. The hypotheses of Corollary 2.1 imply the characteristic conditions stated by Proposition 2.2.

The $-compatibility hypothesis of Corollary 2.1 also has the following meaning. A family {Xα } of Poisson infinitesimal automorphisms has an associated generalized distribution D(Xα ) spanned by the $-Hamiltonian vector fields of the functions f ∈ C ∞ (M) that are constant along the orbits of the vector fields Xα , and this distribution is involutive. span{Xα |N } is a $-compatible normal bundle of N iff D(Xα ) ⊆ T N. If the family {Xα } reduces to one Hamiltonian vector field Xh$ , we have no submanifolds N as in Corollary 2.1 since N should be both tangent and normal to Xh$ . However, we may have the required type of submanifolds if the family consists of a single infinitesimal automorphism X that is not a Hamiltonian vector field. For instance, if D(X) is a regular distribution, it must be a foliation and the leaves of this foliation are Dirac hypersurfaces of M. Before going on with the discussion of Dirac submanifolds, let us also consider some of the situations mentioned at the end of Section 1. Definition 2.2. A normalized submanifold (N, νN ) of the Poisson manifold (M, $) will be called an algebraically Poisson-compatible (a.P.c.) submanifold, respectively, a quasi-Dirac submanifold, if the Poisson bivector field $ is algebraically compatible, respectively, quasi-soldered, to the submanifold. Thus the a.P.c. property is characterized by condition (i) of Definition 2.1, respectively, by the local condition (24), and the quasi-Dirac property is characterized by the local condition (25). The a.P.c. and Dirac properties of a submanifold may hold for more than one normal bundle [10]. A second normal bundle ν˜ N may be defined by (7), and the corresponding local expression of the Poisson bivector field is obtained by switching to the bases (Xa , ∂/∂y u ) in (23). Accordingly, for ν˜ N , the a.P.c. condition is equivalent to ($ab θbu )|N = 0 ⇔ ψ ◦ ($ |ann(T N ) ) = 0, (27) and condition (ii) of Definition 2.1 is equivalent to Xc [$ab θau θbv − $au θav + $av θau + $uv ]|x c =0 = 0. In view of (24), (25), and (27), (28) becomes

(28)


∂$ab u v ∂$av u ∂$ua v ∂$uv w θ θ + θ − θ − θ ∂x c a b ∂x c b ∂x c a ∂y w c

611

x c =0

= 0.

(29)

Condition (27) shows that if $ |ann(T N ) is a surjection, therefore, an isomorphism onto νN (equivalently, det ($ab ) = 0), then νN = $ (ann(νN )) provides the only normalization which makes N an a.P.c. submanifold of M. The submanifolds N such that $ (ann(νN )) is a complement of T N in T M|N are called cosymplectic submanifolds, and it is known that they are Dirac submanifolds [10]. Indeed, the a.P.c. property follows from the skew symmetry of $, and (25) follows from the following component of the Poisson condition [$, $] = 0 in the local adapted coordinates of (23) [8]: ∂$uv [$, $]auv |x c =0 = 2 $ab = 0. (30) ∂x b x c =0 The following result is, obviously, important. Proposition 2.3. If N is either an a.P.c. or a quasi-Dirac submanifold, the bivector field $ = pT ($|N ) is a Poisson bivector field on N . Moreover, in the a.P.c. case, $ does not depend on the choice of the normal bundle among those which satisfy Definition 2.2. Proof. From (23), it follows that 1 ∂ uv ∂ ∧ . $ = $ 2 ∂y u ∂y v x c =0

(31)

Then from [$, $] = 0 and either (24) or (25), we get ⎞ ⎛ u2 u3 ∂$ ⎠ [$, $]u1 u2 u3 |x c =0 = 2 ⎝ $u1 w ∂y w Cycl(u1 ,u2 ,u3 )

= [$ , $ ]u1 u2 u3 = 0;

(32)

x c =0

i.e., $ is a Poisson bivector field on N. Finally, (24) shows that ι∗ ($ (dy u )) = $ (dy u ) (ι : N ⊆ M), and this proves the last assertion.

The Poisson structure $ is said to be induced by the Poisson structure $, and was defined and studied for Dirac submanifolds in [10]. In the a.P.c. case, the submanifold has a second fundamental form (LX $)|ann(νN ) , which vanishes iff N is a Dirac submanifold. Remark 2.1. Several authors have studied a generalization of Poisson structures that consists of a pair ($, ), where $ is a bivector field and is a closed, differential 3-form on the manifold M, such that [$, $] = $ .

(33)

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Such a pair is called a twisted Poisson structure. For details, see [7] and the references of that paper. The notions of an algebraically compatible, a quasi-Dirac and a Dirac submanifold may be defined for twisted Poisson manifolds by asking the bivector field $ to satisfy the same conditions as in the Poisson case. Then the proof of Proposition 2.3 shows that if ι : N → M is a submanifold of one of these three categories, ($ , ι∗ ) is an induced twisted Poisson structure. If σ : W → N is a compatible tubular neighborhood of (N, νN ), the induced Poisson structure is characterized by {f, g}$ = {f ◦ σ, g ◦ σ }$ ◦ ι

(34)

∀f, g ∈ C ∞ (N ) and ι : N ⊆ M. With the same tubular neighborhood, the a.P.c. property is equivalent to the fact that ∀f ∈ C ∞ (N ), the $-Hamiltonian vector field of f ◦ σ is tangent to N or that one has ι∗ ◦ $ = $ ◦ σ ∗ .

(35)

Furthermore, N is a Dirac submanifold if, besides the above, it also has the property that ∀x ∈ N, ∀X ∈ Tx (Wx ), ∀f, g ∈ C ∞ (N ), one has X{f ◦ σ, g ◦ σ }$ = 0.

(36)

We summarize the above remarks in the following. Proposition 2.4. A submanifold N of the Poisson manifold (M, $) is an a.P.c. submanifold iff N is endowed with a Poisson structure $ and has a tubular neighborhood σ : W → N such that conditions (34) and (35) hold. Furthermore, N is a Dirac submanifold iff it is a.P.c. and condition (36) holds, too. Remark 2.2. In [10] the author uses the independence of the induced Poisson structure on the choice of the normal bundle to define local Dirac submanifolds [10] as submanifolds N of the Poisson manifold (M, $) such that ∀x ∈ N , there exists an open neighborhood U in M where N ∩ U is a Dirac submanifold. Proposition 2.3 shows that a local Dirac submanifold also inherits a well-defined, global, induced Poisson structure. In fact, Proposition 2.3 shows that local a.P.c. submanifolds may be defined similarly. Remark 2.3. Proposition 2.4 suggests considering submanifolds N of (M, $) which come endowed with a Poisson structure $ such that for some tubular neighborhood σ : W → N, σ is a Poisson mapping or, equivalently, the brackets {f ◦ σ, g ◦ σ }|$ , which are defined on W , are constant along the fibers of σ . Such submanifolds deserve the name of strong Dirac submanifolds. Obviously, they are Dirac submanifolds, and, with respect to adapted coordinates, one must have ∂$uv /∂x a ≡ 0. The complete lift of the Poisson bivector field $ is a Poisson structure $C called the tangent Poisson structure of $. The tangent structure is exactly the one induced by the Lie algebroid structure of T ∗ M defined by $ on the total space of its dual vector bundle T M. From Proposition 1.3, we get the following characteristic property of Dirac submanifolds.


613

Proposition 2.5 ([10]). The submanifold N of (M, $) is a Dirac submanifold iff there exists a normal bundle νN which is a coisotropic submanifold of (T M, $C ). The following result is significant for the next section. Recall that a Poisson structure $ is homogeneous if there exists a vector field Z ∈ T M such that LZ $ = −$.

(37)

Proposition 2.6. Let N be an a.P.c. submanifold of the homogeneous Poisson manifold (M, $, Z) such that Z|N ∈ T N . Then (N, $ , Z|N ), where $ is the induced Poison structure, also is a homogeneous Poisson manifold. Proof. If the homogeneity condition (37) is evaluated on (dϕ, dψ) (ϕ, ψ ∈ C ∞ (M)), one gets the equivalent condition $ {ϕ, ψ}$ = Z{ϕ, ψ}$ − [Z, Xϕ$ ]ψ + [Z, Xψ ]ϕ,

(38)

where X denotes Hamiltonian vector fields. Now let σ : W → N be a tubular neighborhood of N where the conditions of Proposition 2.4 hold. Then (38), written for ϕ = f ◦ σ , ψ = g ◦ σ (f, g ∈ C ∞ (M)) and composed by ι, provides the similar condition (38) for $ .

Now we point out the existence of a specific cohomology related with a Dirac submanifold (N, νN ) of the Poisson manifold (M, $). Namely, since the Poisson bivector field $ is soldered to N , V(M, N, νN) = (V k (M, N, νN), ∂$ = −[$, .])

(39)

is a subcomplex of the Lichnerowicz–Poisson cochain complex of (M, $) (e.g., [8]); k (M, N, νN) that will be called soldered therefore, it defines cohomology spaces HsP Poisson cohomology spaces. Proposition 2.7. The homomorphism $ : T ∗ M → T M induces homomorphisms k k k$ : HsdeR (M, N, νN) −→ HsP (M, N, νN).

(40)

If the Poisson structure $ is defined by a symplectic form ω, the mappings (40) are isomorphisms. Proof. Using adapted local coordinates, it is easy to check that ∀κ ∈ k (M, N, νN), $ κ ∈ V k (M, N, νN) and, as for the general Poisson cohomology, ∂$ ◦$ = −$ ◦d. This justifies the existence of the homomorphisms (40). In the symplectic case, N must be a symplectic (2n)-dimensional submanifold of (M 2m , ω), and νN must be the ω-orthogonal bundle of T N [10]. Indeed, each ∗ ∗ point x ∈ N has an open neighborhood with coordinates (x a , x a , y u , y u ) (a = 1, . . . , m − n, u = 2m − 2n + 1, . . . , 2m − n, a ∗ = a + m − n, u∗ = u + n) such that ∗ ∗ ω= dx a ∧ dx a + dy u ∧ dy u , (41) a

u

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and N has the local equations x a = 0, x a = 0 [6]. Obviously, these coordinates also are adapted coordinates with respect to the ω-orthogonal bundle νN of T N. The uniqueness of the normal bundle follows from (27). Then $ has the inverse −0ω , and the latter induces the inverses of the homomorphisms (40).

We end this section by a brief discussion of the same subject in Nambu–Poisson geometry. A Nambu–Poisson manifold of order k is a manifold M m endowed with a Nambu–Poisson tensor field , i.e., a k-vector field Q ∈ V k (M) (k ≥ 3) which, when evaluated on differentials, defines a skew-symmetric bracket of k functions {f1 , . . . , fk } = Q(df1 , . . . , dfk ) that satisfies the generalized Jacobi identity {f1 , . . . , fk−1 , {g1 , . . . , gk }} =

k

(42)

{g1 , . . . , gh−1 , {f1 , . . . , fk−1 , gh }, gh+1 , . . . , gk }.

h=1

It is known that Q is a Nambu–Poisson tensor field iff it is decomposable (i.e., a wedge product of k vectors) at each point, and its components in every local chart satisfy the equality ( ) m k i1 ...ik−1 h j1 ...jk j1 ...jl−1 hjl+1 ...jn i1 ...ik−1 jl Q . (43) ∂h Q − Q ∂h Q h=1

l=1

Another basic result tells that around each point x ∈ M where Qx = 0, there are local coordinates such that Q=

∂ ∂ ∧ ··· ∧ k ∂x ∂x 1

(44)

(e.g., see [9] for details). Accordingly, it is natural to define the following. Definition 2.3. Let (M m , Q) be a Nambu–Poisson manifold of order k and (N n , νN) (n ≥ k) a normalized submanifold. Then N is an algebraically compatible, a quasiDirac, or a Dirac submanifold if Q is algebraically compatible, quasi-soldered or soldered, respectively, to N. Obviously, the projection Q = pT (Q|N ) is a decomposable k-vector field on N. Then a straightforward examination of condition (43), where the components of Q are as in formula (17), and an argument similar to that at the end of the proof of Proposition 2.3 show that we have the following. Proposition 2.8. If (N, νN ) is either an algebraically compatible or a quasi-Dirac (Dirac) submanifold of the Nambu–Poisson manifold (M, Q) of order k, Q is an induced Nambu–Poisson k-vector field on N . Moreover, if algebraic compatibility holds, Q does not depend on the choice of νN .


615

Example 2.1. Consider the Nambu–Poisson manifold (Rm , Q), where Q is globally defined by (44) with the canonical coordinates of Rm . Let N n (n ≥ k) be the ndimensional plane defined by the equations x n+s =

n

cun+s x u + p n+s ,

s = 1, . . . , m − n,

(45)

u=1

where cun+s , pn+s = const. Then the tangent spaces of N are spanned by the vector fields m−n ∂ ∂ Xu = u + cun+s n+s , u = 1, . . . , n, ∂x ∂x s=1

and we may define a normalization where the normal bundle νN is spanned by (∂/∂x n+s )m−n s=1 . It follows easily that with this normalization, N is a quasi-Dirac submanifold with the induced Nambu–Poison structure Q = X1 ∧ · · · ∧ Xk . Furthermore, (N, νN ) above is a Dirac submanifold iff cun+s = 0 for u = 1, . . . , k; s = 1, . . . , m − n. In the Nambu–Poisson case, we may also distinguish a situation similar to that of the cosymplectic submanifolds of a Poisson manifold. Indeed, the interior product by a (k − 1)-form defines a vector bundle morphism Q : ∧k−1 T ∗ M → T M and the submanifold N of M will be called cosymplectic if im(Q |ann(T N )⊗∧k−2 T ∗ M ) is a normal bundle νN of the submanifold N . Then we get the following. Proposition 2.9. Any cosymplectic submanifold N n (n ≥ k) of a Nambu–Poisson manifold (M, Q) of order k is a Dirac submanifold. Proof. Of course, the normalization we have in mind is that produced by the definition of a cosymplectic submanifold, i.e., νN is spanned by the vector fields i(dx a ∧ dy u1 ∧ · · · ∧ dy uk−2 )Q = (−1)k−1 Qbau1 ...uk−2 + Qau1 ...uk−2 v

∂ ∂x b

(46)

∂ , ∂y v

where the local coordinates and components are those of the formula (17). The normality of these vectors implies that Q satisfies the condition of algebraic compatibility Qau1 ...uk−2 v = 0. The condition of cosymplecticity means that there are m−n choices of the group of indices (a, u1 , . . . , uk−2 ) with linearly independent corresponding vector fields (46). Then (43) written for these choices of the indices implies the fact that Q is quasi-soldered to (N, νN ).

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3 Dirac submanifolds of Jacobi manifolds For a detailed study of Jacobi manifolds we refer the reader to [1] and its references. Jacobi manifolds are a natural generalization of Poisson manifolds namely, a Jacobi structure on a manifold M m is a Lie algebra bracket {f, g} on C ∞ (M), which is given by bidifferential operators. It follows that one must have {f, g} = (df, dg) + f Eg − gEf,

(47)

where E is a vector field and is a bivector field on M such that4 [, ] = −2E ∧ ,

LE = 0.

(48)

Thus if E = 0, we have a Poisson structure. The Jacobi structure (M, , E) is equivalent to the homogeneous Poisson structure ∂ ∂ ∧ E), Z= $ = e−τ ( + (49) ∂τ ∂τ on M × R; M will then be identified with M × {0}. For instance [5], let $ be a linear Poisson structure on Rn \{0}, and consider the diffeomorphism S n−1 × R ≈ Rn \{0} defined by n x i = e−τ ui , (ui )2 = 1, τ ∈ R. i=1

Then it is easy to check that $ must be of the form (49), which provides a Jacobi structure on S n−1 . We call this structure a Lichnerowicz–Jacobi structure of the sphere. On a Jacobi manifold, one may define Hamiltonian vector fields Xf = df + f E

(f ∈ C ∞ (M)),

(50)

and they span a generalized foliation S such that the leaves of S are either contact or locally conformal symplectic manifolds. For instance, in the case of a Lichnerowicz– Jacobi structure the leaves are the orbits of the quotient coadjoint representation of a connected Lie group G with the Lie algebra G of structure constants defined by the corresponding linear Poisson structure $ (see above), i.e., the action defined on S n−1 by the coadjoint action of G on G ∗ \{0} ≈ Rn \{0} if S n−1 is seen as a quotient space of G ∗ \{0} [5]. Another important fact we want to recall is that ∀ϕ ∈ C ∞ (M), the bracket {f, g}ϕ = e−ϕ {eϕ f, eϕ g}

(51)

is a Jacobi bracket said to have been obtained by a conformal change of the original bracket. The tensor fields of the new bracket are ϕ = eϕ ,

E ϕ = eϕ (E + i(dϕ)).

(52)

Now we begin our considerations on submanifolds. 4 The minus sign comes from our sign convention for the Schouten–Nijenhuis bracket in

Section 1.


617

Definition 3.1. Let (N, νN ) be a normalized submanifold of the Jacobi manifold (M, , E). Then (1) N is an almost Dirac submanifold if is an N -soldered bivector field; (2) N is an algebraically Jacobi-compatible (a.J.c.) submanifold if and E are algebraically compatible with the normalization of N ; (3) N is a (quasi-)Dirac submanifold if and E are (quasi-)soldered to (N, νN ). Equivalently, N is an almost Dirac submanifold if each point x ∈ N has a neighborhood with adapted coordinates as in Section 1 such that =

1 ab ∂ ∂ ∂ ∂ ∂ 1 ∂ ∧ + au a ∧ u + uv u ∧ v , 2 ∂x a ∂x b ∂x ∂y 2 ∂y ∂y

(53)

where au |x c =0 = 0, ∂uv = 0. ∂x a c

(54) (55)

x =0

Then N is a Dirac submanifold if, furthermore, the vector field E is tangent to N and has the local expression ∂ ∂ E = a a + u u , (56) ∂x ∂y where ∂ u = 0. (57) a |x c =0 = 0, ∂x a x c =0 For the quasi-Dirac case, we only have the condition (55) and the second equality (57). Finally, N is an a.J.c. submanifold if (54) and the first condition (57) hold. Proposition 3.1. Let (N, νN ) be either an almost Dirac or an a.J.c. or a quasiDirac submanifold of the Jacobi manifold (M, , E). Then [ = pT (|N ), E = pT (E|N )] is a Jacobi structure on N . Furthermore, in the almost Dirac and the a.J.c. case does not depend on the choice of the normalization. Proof. With local adapted coordinates, we have 1 ∂ ∂ = uv u ∧ v 2 ∂y ∂y x c =0

(58)

and ⎛ [, ]u1 u2 u3 |x c =0 = 2 ⎝

u1 a

Cycl(u1 ,u2 ,u3 )

+

Cycl(u1 ,u2 ,u3 )

∂u2 u3 ∂x a

(59)

⎞ u2 u3 ∂ ⎠ u1 w ∂y w

x c =0

= [ , ]u1 u2 u3 .

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Hence in all the cases of the proposition, we have [ , ] = pT ([, ]|N ) = −2E ∧ . Then an examination of the coordinate expression of LE , where E and are given by (56) and (53), respectively, shows that the conditions (54) and (55), as well as either (54) and the first condition (57) or (55) and the second condition (57), imply that LE = pT (LE |N ) = 0. Finally, where asserted, the independence of of the normalization follows from

ι∗ ( (dy u ) = (dy u ), ι : N ⊆ M. We notice that formula (59) also implies the following. Proposition 3.2. Let (N, νN ) be a normalized submanifold of the Jacobi manifold (M, , E) such that is algebraically compatible with the normalization and E is a normal field of N. Then is a Poisson structure on N , and it is independent on the choice of νN among all possible choices that contain E|N . The Jacobi or Poisson structures defined on N by ( , E ) are said to be induced by (, E). In the cases where only algebraic compatibility holds, invariants of the second fundamental form type (LX )|ann(νN ) , [X, E]|ann(νN ) , where X is normal to N, appear. Proposition 1.2 allows us to give some simple examples. Consider the Jacobi manifold M = R3n+1 with ⎞ ⎛ n n ∂ ∂ ∂ ∂ ∂ ⎠, E=t (60) ui i ∧ + t pj = ∧⎝ ∂q ∂pi ∂t ∂pj ∂t i=1

j =1

(the variables of (60) are the natural coordinates of M). Then the hyperplane t = 0 is the fixed point locus of the involution (ui , q i , pi , t) → (ui , q i , pi , −t). This involution preserves the tensor fields (60); hence the hyperplane t = 0 is a Dirac submanifold with an induced Poisson structure. For the same M, the involution (ui , q i , pi , t) → (−ui , −q i , pi , t) also preserves (60); hence its fixed point locus, which is the (n + 1)-plane ui = 0, q i = 0, is a Dirac submanifold with an induced Jacobi structure. Finally, if we restrict M to the domain pi > 0, t > 0 and consider the involution that sends t to 1/t and preserves the other coordinates, only of (60) is preserved hence, the fixed point locus, which is the hyperplane t = 1, is an almost Dirac submanifold. Moreover, the last involution sends E to −E. Therefore, E is normal to the submanifold, and the induced structure is a Poisson structure. Another interesting fact is the following. Proposition 3.3. Let (M, , E) be a Jacobi manifold, and (M × R, $), with $ defined by (49), the corresponding homogeneous Poisson manifold. Then N is an a.J.c. or a Dirac submanifold of the former iff N × R is an a.P.c., respectively, Dirac, submanifold of the latter.


619

Proof. We will use the lift of νN to N ×R as a normal bundle. τ of (49) is a coordinate along N × R, and we see that if and E are of the local form (53), (56) then $ satisfies the conditions (24), (25), and conversely.

From Proposition 1.3 it follows that the almost Dirac and Dirac submanifolds of a Jacobi manifold may also be characterized by using the tangent bundle T M; namely, we have the following. Proposition 3.4. The normalized submanifold (N, νN ) is almost Dirac iff the submanifold νN of T M is such that C (ann(T νN )) ⊆ T νN , where C is the complete lift of . Furthermore, N is a Dirac submanifold iff besides the previous condition, one also has E C ∈ (T νN), where E C is the complete lift of the vector field E. Remark 3.1. The tensor fields (C , E C ) do not define a Jacobi structure on T M. A tangent Jacobi structure can be obtained by considering the Poisson structure induced on the manifold T M × R by the Lie algebroid J 1 M = T ∗ M × R of (, E) [4]. Namely, with the notation of (20), (21), if we associate with each cross-section (f, αi dzi ) ∈ J 1 M the function eτ (f + αi z˙ i ) ∈ C ∞ (T M × R), the Lie algebroid bracket of J 1 M yields a Poisson bracket of the specified kind of functions, which extends to a Poisson bracket on C ∞ (T M × R). Computations show that the Poisson bivector of this structure is 4 5 ∂ ˜ = e−τ C − V − E ∧ (E C − E V ) + $ ∧ EC , (61) ∂τ where the upper index V denotes the vertical lift [11] and E is the Euler vector field , i.e., EV = Ei

∂ , ∂ z˙ i

V =

1 ij ∂ ∂ ∧ j, i 2 ∂ z˙ ∂ z˙

E = z˙ i

∂ . ∂ z˙ i

(62)

Accordingly, (C − V − E ∧ (E C − E V ), E C ) is a Jacobi structure on T M, which deserves the name of tangent Jacobi structure. A particular class of Dirac submanifolds was studied in [1], and here we reprove the following. Proposition 3.5 ([1]). Assume that N is a submanifold of (M, , E) such that (ann(T N )) is a normal bundle νN of N. Then N is a Dirac submanifold iff the vector field E is tangent to N . Furthermore, there always exists a conformal change (51), with ϕ|N = 0, such that N is a Dirac submanifold of (M, ϕ , E ϕ ). Proof. If N is a Dirac submanifold, E ∈ T N by definition. For the converse, we use the normal bundle of the hypothesis, and represent and E by (53) and (56), respectively. Clearly, the choice of νN is such that (dx a ) ∈ νN along N , which is equivalent to (54). If this condition holds, the auv-component of the first equality (48) yields

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ab ∂

uv

∂x b

+E a

uv

|N = 0.

(63)

Since (ann(T N )) is normal to N iff the matrix (ab ) is nondegenerate, we see that E tangent to N implies (55). Furthermore, if E|N ∈ T N , the second equality (48) yields ∂E u ab b = 0; (64) ∂x N therefore, (57) holds. Concerning the last part of the proposition, (52) shows that the required conformal transformation exists if there exists a function ϕ ∈ C ∞ (M), which vanishes on N and is such that ∂ϕ E a |N = ab b . (65) ∂x N Since (ab ) is nondegenerate, the conditions for ϕ prescribe the 1-jet with respect to the variables (x a ) of ϕ at the points of N . Therefore, a required function ϕ exists around every point of N . Then these local solutions may be glued up by a partition of unity along N. (See also the argument of [1].)

We end by a discussion of Dirac submanifolds of the transitive Jacobi manifolds, i.e., locally conformal symplectic (l.c.s.) and contact manifolds [1]. Proposition 3.6. A submanifold N is an almost Dirac submanifold of the l.c.s. manifold M iff it is Dirac, and this happens iff N inherits from M an induced l.c.s. structure. Moreover, there is only one possible normal bundle, the symplectic orthogonal bundle of T N. Proof. Recall that the l.c.s. structure of M is a nondegenerate 2-form such that for some open covering M = ∪α Uα , ∀α |Uα = e−σα α , where σα are functions, α are 2-forms and d α = 0. Equivalently, d = ω ∧ , where ω is the closed 1-form defined by gluing up the local forms dσα (ω is called the Lee form). It is known that M is a Jacobi manifold with the structure defined by the bivector field , where = 0−1

, and the vector field E = ω [1]. Assume that N is an almost Dirac submanifold with the normal bundle νN . Then |ann(T N ) is an isomorphism onto νN, which, as in (27), ensures the uniqueness of νN , and |ann(νN ) is an isomorphism on T N, which is equivalent to the fact that ι∗ (ι : N ⊆ M) is nondegenerate and provides an l.c.s. structure on N . Accordingly, we may use Marle’s theorem [6], and find local coordinates of N on some neighborhood Uα such that with the notation of (41), one has ' * ∗ ∗ (66)

|Uα = e−σα dx a ∧ dx a + dy u ∧ dy u . a

u

Obviously, this expression of implies that νN is -orthogonal to T N and that the coordinates used in (66) are adapted coordinates.


621

Now condition (55) applied to (66) becomes (∂σα /∂x a )x c =0 = 0, i.e., ωa |x c =0 = 0. Furthermore, one of the conditions that express dω = 0 is ∂ωa /∂y u = ∂ωu /∂x a , whence we also get (∂ωu /∂x a )x c =0 = 0. Therefore, the Lee form ω, and the vector field E too, are soldered to N , and N must be a Dirac submanifold of M. The converse part of the proposition follows from (66).

Proposition 3.7. Let M 2m+1 be a contact manifold with the contact 1-form θ. Then a submanifold ι : N ⊆ M is a Dirac submanifold iff ι∗ θ is a contact form on N. Furthermore, the normal bundle of N is unique, and it is the dθ -orthogonal bundle of T N. Proof. Recall that θ is a contact form iff θ ∧ (dθ )m vanishes nowhere. A contact form produces a Jacobi structure [1], which consists of the vector field E defined by i(E)θ = 1,

i(E)dθ = 0,

(67)

and the bivector field (df, dg) = dθ(Xfθ , Xgθ )

(f, g ∈ C ∞ (M)),

(68)

where the Hamiltonian vector field Xfθ is defined by i(Xfθ )θ = f,

i(Xfθ )dθ = −df + (Ef )θ.

(69)

From (69) we get Xfθ = df + f E,

(df, dg) = dθ ( df, dg).

(70)

If M is the contact manifold above, M × R has the Poisson bivector $ given by (49), and it also has the symplectic form

= eτ (dθ + dτ ∧ θ ).

(71)

An easy computation shows that all the functions of the form eτ f ∈ C ∞ (M × R) (τ ∈ R, f ∈ C ∞ (M)) have the same Hamiltonian vector fields with respect to $ and . Therefore, $ ◦ 0 = − Id . Now Proposition 3.3 states that N is a Dirac submanifold of M iff N ×R is a Dirac submanifold of M × R. In the present case, this means that N × R is a symplectic submanifold of (M × R, ), and it follows that (N, ι∗ θ ) must be a contact manifold, and that the normal bundle must be the one indicated by the proposition.

References [1] P. Dazord, A. Lichnerowicz, and Ch.-M. Marle, Structure locale des variétés de Jacobi, J. Math. Pure Appl., 70 (1991), 101–152. [2] I. Dorfman, Dirac Structures and Integrability of Nonlinear Evolution Equations, Wiley, New York, 1993.

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[3] J. Huebschmann, Lie-Reinhart algebras, Gerstenhaber algebras and Batalin-Vilkoviski algebras, Ann. Inst. Fourier (Grenoble), 48 (1998), 425–440. [4] Y. Kerbrat and Z. Souici-Benhammadi, Variétés de Jacobi et groupoïdes de contact, C. R. Acad. Sci. Paris Sér. I Math., 317 (1993), 81–86. [5] A. Lichnerowicz, Représentation coadjointe quotient et espaces homogènes de contact ou localement conformément symplectiques, J. Math. Pures Appl., 65 (1986), 193–224. [6] Ch.-M. Marle, Sous-variétés de rang constant d’une variété symplectique, Astérisque, 107–108 (1983), 69–86. [7] P. Ševera and A. Weinstein, Poisson geometry with a 3-form background, Progr. Theorer. Phys. Suppl., 144 (2001), 145–154. [8] I. Vaisman, Lectures on the Geometry of Poisson Manifolds, Progress in Mathematics, Vol. 118, Birkhäuser, Basel, 1994. [9] I. Vaisman, A survey on Nambu-Poisson brackets, Acta Math. Univ. Comenianae, 68 (1999), 213–241. [10] P. Xu, Dirac submanifolds and Poisson involutions, Ann. Sci. Ec. Norm. Sup., 36 (2003), 403–430. [11] K. Yano and S. Ishihara, Tangent and Cotangent Bundles, Marcel Dekker, New York, 1973.

Quantum maps and automorphisms∗ Steve Zelditch Department of Mathematics Johns Hopkins University Baltimore, MD 21218 USA [email protected] Abstract. There are several inequivalent definitions of what it means to quantize a symplectic map on a symplectic manifold (M, ω). One definition is that the quantization is an automorphism of a ∗-algebra associated to (M, ω). Another is that it is unitary operator Uχ on a Hilbert space associated to (M, ω), such that A → Uχ∗ AUχ defines an automorphism of the algebra of observables. A yet stronger one, common in partial differential equations, is that Uχ should be a Fourier integral operator associated to the graph of χ. We compare the definitions in the case where (M, ω) is a compact Kähler manifold. The main result is a Toeplitz analogue of the Duistermaat–Singer theorem on automorphisms of pseudodifferential algebras, and an extension which does not assume H 1 (M, C) = {0}. We illustrate with examples from quantum maps.

1 Introduction Much attention has been focussed recently on ∗ products on Poisson manifolds (M, {, }) (see, among others, [Kontsevich (1997)], [Cattaneo–Felder (2000)], [Karabegov–Schlichenmaier (2001)], [Tamarkin (1998)], [Reshetikhin–Takhtajan (1999)], [Etingof–Kazhdan (1996)], [Weinstein–Xu (1998)], [Boutet de Monvel 5 (2002)]). Such ∗ products are viewed as quantizing functions on M to an algebra of observables, which we will refer to as a ∗ product algebra, or more simply as a ∗-algebra. This article is concerned with the related problem of quantizing symplectic maps χ on Kähler manifolds (M, ω), a special case of the problem of quantizing Poisson maps. From the ∗-algebra viewpoint, it seems most natural to quantize such a symplectic map as an automorphism of a ∗-algebra associated with (M, ω), specifically the (complete) symbol algebra T ∗ /T −∞ of Berezin–Toeplitz operators over (M, ω). These symbol algebras are basic examples of abstract ∗-algebras arising in deformation quantization of Poisson manifolds (see [Boutet de Monvel 1 (1999)], [Boutet de Monvel 3 (1999)], [Boutet de Monvel 5 (2002)], [Charles (2003)], [Cattaneo–Felder (2000)], [Guillemin (1995)], [Schlichenmaier (1999)], [Schlichenmaier ∗ This research was partially supported by NSF grant DMS-0071358 and by the Clay Math-

ematics Institute.

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(1998)] for more on this aspect). But they carry more structure than bare ∗-algebras: the Toeplitz operator algebra T ∗ of which T ∗ /T −∞ is the symbol algebra also comes with a representation as operators on a Hilbert space. In the Hilbert space setting, it is most natural to try to quantize a symplectic map χ as a unitary operator Uχ , and to induce the automorphism Uχ AUχ∗ on T ∗ . As will be explained below (see also [Zelditch (1997)]), it is not always possible to quantize a symplectic map this way. When possible, the quantization Uχ is an example of what is known as a quantum map in the literature of quantum chaos. Such quantum maps have also been the focus of much attention in recent years by a virtually disjoint group (see, e.g., [de Biévre–degli Esposti (1998)], [Keating (1991)], [degli Esposti–Graffi–Isola (1995)], [Hannay–Berry (1980)], [Marklof–Rudnick (2000)], [Zelditch (1997)]). The main purpose of this article is to contrast the different notions of quantizing symplectic maps, as as they arise in Toeplitz ∗-algebras, partial differential equations and quantum chaos. Aside from its intrinsic interest, the relation between quantum maps and automorphisms of ∗-algebras has practical consequences in quantum chaos, i.e., in the relations between dynamical properties of χ and the eigenvalues/eigenfunctions of its quantization Uχ . In the physics literature of quantum chaos, quantum maps are studied through examples such as quantum kicked tops (on S 2 ), cat maps, rotors, baker’s map and standard maps (on the 2-torus T2 ). Almost always, the quantizations are given as explicit unitary matrices UN (depending on a Planck constant 1/N ) on special Hilbert spaces HN , often using some special representation theory, and no formal definition is given of the term “quantum map.’’The need for precise definitions is felt, however, as soon as one aims at quantizing maps which lie outside the range of standard examples. Even symplectic maps on surfaces of genus g ≥ 2 count as nonstandard, and only seem to have been quantized by the Toeplitz method discussed in this paper and in [Zelditch (1997)]. A further reason to study quantum maps versus automorphisms is to better understand obstructions to quantizations. It is often said that Kronecker translations Tα,β (x, ξ ) = (x + α, ξ + β),

(x, ξ ) ∈ R2n /Z2n

and affine symplectic torus maps fα (x, ξ ) = (x + ξ, ξ + α) are not quantizable, for reasons explained in Proposition 2.2. Nevertheless, the paper [Marklof–Rudnick (2000)] proposes a quantization of such maps. Of course, the resolution of this paradox is that a weaker notion of quantization is assumed in [Marklof–Rudnick (2000)] than elsewhere, as will be explained below. The implicit criterion (including that in [Marklof–Rudnick (2000)]) that UN quantize a symplectic map χ is that the Egorov-type formula UN∗ OpN (a)UN ∼ OpN (a ◦ χ )

(N → ∞)

(1)

hold for all elements OpN (a) of the algebra TN of observables, where χ is a symplectic map of (M, ω). Postponing precise definitions, we see that the operative condition is

Quantum maps and automorphisms

625

that UN∗ OpN (a)UN defines an automorphism of TN , at least to leading order. Here, our notation for observables and quantum maps are in terms of sequences as the inverse Planck constant N varies. We temporarily write T ∗ for sequences {OpN (a)} of observables (with T −∞ the sequences which are rapidly decaying in N ), and U ∼ {UN } for sequences of unitary quantum maps. We will soon give more precise definitions. We now distinguish several notions of quantizing a symplectic map and make a number of assertions which will be justified in the remainder of the article. •

•

•

•

•

•

There is a geometric obstruction to quantizing a symplectic map χ as a Toeplitz quantum map Uχ ,N on HN (see Definition 1.5 and Proposition 2.2). Kronecker translations and parabolic maps of the torus are examples of nonquantizable symplectic maps in the Toeplitz sense (see Propositions 5.1 and 5.3). There is no obstruction to quantizing a symplectic map as an automorphism of the Toeplitz symbol algebra T ∗ /T −∞ (see Theorem 1.6). For instance, Kronecker maps and cat maps are quantizable as automorphisms (see Propositions 5.2–5.4). Conversely, if H 1 (M, C) = {0}, then every order-preserving automorphism of the symbol algebra T ∗ /T −∞ on M is induced by a symplectic map of (M, ω) (see Theorem 1.6 for this and for the case where H 1 (M, C) = {0}). There is an obstruction to “extending’’ an automorphism α of T ∗ /T −∞ as an automorphism of T ∗ . In particular, there is an obstruction to inducing automorphisms αN of the finite-dimensional algebras of operators TN acting on HN (see Theorem 1.6). Again, Kronecker maps are examples (see Section 5). Any sequence UN of unitaries on HN which defines an automorphism of T ∗ /T −∞ must be a Toeplitz quantum map in sense of Definition 1.5(i) (see [Boutet de Monvel 4 (1985)], [Zelditch (1997)]). Many of the key problems of quantum chaos, e.g., problems on eigenvalue level spacings or pair correlation, on ergodicity and mixing of eigenfunctions (etc.) concern only the spectral theory of the automorphism quantizing χ and not the unitary map per se (see Section 6).

1.1 The Toeplitz setup In order to state our results precisely, we need to specify the framework in which we are working. The framework of Toeplitz operators used in this paper is the same as in [Boutet de Monvel 1 (1999)], [Boutet de Monvel 2 (1998)], [Guillemin (1995)], [Bleher–Shiffman–Zelditch (2001)], [Shiffman–Zelditch], [Zelditch (1997)], [Zelditch (1998)]. We briefly recall the notation and terminology. Our setting consists of a compact, connected Kähler manifold (M, ω) with 1 [ω] ∈ H 1 (M, Z). Under this integrality condition, there exists a positive Her2π mitian holomorphic line bundle (L, h) → M over M with curvature form √ −1 ¯ ∂ ∂ log eL h = ω, c1 (h) = − π where eL is a nonvanishing local holomorphic section of L, and where eL h = 1 m h(eL , eL )1/2 denotes the h-norm of eL . We give M the volume form dV = m! ω .

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The Hilbert spaces “quantizing’’ (M, ω) are then defined to be the spaces H 0 (M, LN ) of holomorphic sections of LN = L ⊗ · · · ⊗ L. The metric h induces 0 N Hermitian metrics hN on LN given by s ⊗N hN = sN h . We give H (M, L ) the inner product s1 , s2 = hN (s1 , s2 )dV (s1 , s2 ∈ H 0 (M, LN )), (2) M

and we write |s| = s, s1/2 . We then define the Szegö kernels as the orthogonal projections $N : L2 (M, LN ) → H 0 (M, LN ), so that ($N s)(w) = hN s ∈ L2 (M, LN ). (3) z (s(z), $N (z, w))dVM (z), M

Instead of dealing with sequences of Hilbert spaces, observables and unitary operators, it is convenient to lift them to the circle bundle X = {λ ∈ L∗ : λh∗ = 1}, where L∗ is the dual line bundle to L, and where h∗ is the norm on L∗ dual to h. ¯ X and the volume form Associated to X is the contact form α = −i∂ρ|X = i ∂ρ| dVX =

1 α ∧ (dα)m = α ∧ π ∗ dVM . m!

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Holomorphic sections then lift to elements of the Hardy space H2 (X) ⊂ L2 (X) of square-integrable CR functions on X, i.e., functions that are annihilated by the Cauchy–Riemann operator ∂¯b and are L2 with respect to the inner product 1 F1 , F2 = F1 F2 dVX , F1 , F2 ∈ L2 (X). (5) 2π X We let rθ x = eiθ x (x ∈ X) denote the S 1 action on X and denote its infinitesimal genO ∂ 2 (X), erator by ∂θ . The S 1 action on X commutes with ∂¯b ; hence H2 (X) = ∞ H N =0 N 2 (X) = {F ∈ H2 (X) : F (r x) = eiN θ F (x)}. A section s of LN deterwhere HN θ N mines an equivariant function sˆN on L∗ by the rule sˆN (λ) = (λ⊗N , sN (z)),

λ ∈ L∗z ,

z ∈ M,

where λ⊗N = λ⊗· · ·⊗λ. We henceforth restrict sˆ to X and then the equivariance property takes the form sˆN (rθ x) = eiN θ sˆN (x). The map s → sˆ is a unitary equivalence 2 (X). We refer to [Boutet de Monvel–Guillemin (1981)], between H 0 (M, LN ) and HN [Boutet de Monvel–Sjöstrand (1976)], [Bleher–Shiffman–Zelditch (2001)], [Zelditch (1998)] for further background. We now define the (lifted) Szegö kernel of degree N to be the orthogonal projection 2 (X). It is defined by $N : L2 (X) → HN $N F (x) = $N (x, y)F (y)dVX (y), F ∈ L2 (X). (6) X

The full Szegö kernel is the direct sum


$=

∞ D

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$N .

N =1

Following Boutet de Monvel–Guillemin [Boutet de Monvel–Guillemin (1981)], we then define the following. Definition 1.1. The ∗-algebra T ∗ (M) of Toeplitz operators of (M, ω) is the algebra of operators on H2 (X) of the form $A$ =

∞ D N =1

$N AN $N , A ∈ #S∗1 (X),

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where #S∗1 (X) is the algebra of pseudodifferential operators of integral order over X which commute with the S 1 action, and where 1 AN = ei N θ Ae−iN θ dθ. (9) 2π S 1 ∂ Here [A, N ] = 0, where N = 1i ∂θ is the operator generating the S 1 action, 2 whose eigenvalue in HN (X) equals N . Since the symbol of A is S 1 -invariant, a Toeplitz operator of order s possesses an expansion ∞ $A$ ∼ N s $aj $N −j , (10) j =0

where aj ∈

C ∞ (M).

We may also express it in the direct sum form $A$ =

∞

$ N aN $ N ,

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N =1 s is a semiclassical symbol of some order s, i.e., admits an where aN (z, z¯ ) ∈ Sscl asymptotic expansion

aN (z, z¯ ) ∼ N s

∞

N −j aj (z, z¯ ),

aj (z, z¯ ) ∈ C ∞ (M)

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j =0

in the sense of symbols. We define the order of a Toeplitz operator $A$ to be the order s of the symbol. The order defines a filtration of T ∗ by spaces of operators T s of order s ∈ Z. See [Guillemin (1995)] for further background. −∞ We also define “flat’’ symbols f (z, N ) ∈ Sscl , denoted f ∼ 0, as functions −m satisfying f = O(N ) for all m. We then define T −∞ to be the flat (or smoothing) Toeplitz operators (possessing a flat symbol). The following definition is important in distinguishing the automorphisms that concern us. Definition 1.2. The complete Toeplitz symbol algebra (or smooth Toeplitz algebra) is the quotient algebra T ∗ /T −∞ .

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O We often view ∞ N =1 $N aN $N as the sequence {$N aN $N } of operators on the sequence HN ! H 0 (M, LN ) of Hilbert spaces. The physicists’ notation for $N aN $N is OpN (aN ). Viewing symbols as sequences {aN (z, z¯ ), we define the ∗N product by $N aN $N ◦ $N bN $N = $N aN ∗N bN $N . (13) In the appendix (Section 7), we will describe the calculation of aN ∗N bN so that it will not seem abstract to the reader. We now introduce automorphisms. Definition 1.3. An order-preserving automorphism α of T ∗ /T −∞ is an automorphism which preserves the filtration T s /T −∞ . We denote the algebra of such automorphisms by Aut o (T ∗ /T −∞ ). It is important to distinguish • •

order-preserving automorphisms of T ∗ that preserve T −∞ ; order-preserving automorphisms of the symbol algebra T ∗ /T −∞ .

Since elements of T ∗ and of T ∗ /T −∞ commute with the S 1 action, either kind of automorphism satisfies * ' ∞ ∞ D D α $ N aN $ N ∼ $ N bN $ N , (14) N =1

N =1

where bN is a semiclassical symbol of the same order as aN . In the case of automorphisms of T ∗ , we can conclude that α($N aN $N ) = $N bN $N and that α induces automorphisms αN of the finite-dimensional algebras TN for fixed N . However, for automorphisms of T ∗ /T −∞ in general, α($N aN $N ) is not even defined since $N aN $N ∈ T −∞ . To put it another way, we cannot uniquely represent an element of the finite-dimensional algebra as $N aN $N although we can uniquely represent elements of T ∗ /T −∞ this way. 1.1.1 Covariant and contravariant symbols Let $N a$N be a Toeplitz operator. By the contravariant symbol of $N aN $N is meant the multiplier aN . By the covariant symbol of an operator F is meant the function F zN , w $N F $N (z, z) N |z=w = , (15) fˆ(z, z¯ ) = zN , w $N (z, z) N where $N (z, w) w (16) N (z) = $N (·, z) is the L2 -normalized “coherent state’’ centered at w. When F = $N a$N , we get a(z, ˆ z¯ ) =

$N a$N (z, z) . $N (z, z)

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We use the notation IN (a) = aˆ for the linear operator (the Berezin transform) which takes the contravariant symbol to the covariant symbol (see [Reshetikhin–Takhtajan (1999)] for background).


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1.2 Statement of results Let us now consider the senses in which we can quantize symplectic maps in our setting. The first sense is that of quantizations of symplectic maps as Toeplitz Fourier integral operators. The definition is as follows. Definition 1.4. Suppose that the symplectic map χ of (M, ω) lifts to (X, α) as a contact transformation χ˜ . By the Toeplitz Fourier integral operator (or quantum map) defined by χ we mean an operator D U= Uχ ,N , Uχ ,N = $N Tχ σN $N , N

where Tχ : L2 (X) → L2 (X) is the translation Tχ (f ) = f ◦ χ˜ −1 and where σN is a symbol designed to make Uχ ,N unitary. (Such a symbol always exists [Zelditch (1997)].) We now distinguish several notions of quantizing a symplectic map. Definition 1.5. Let χ be a symplectic map of (M, ω). In descending strength, we say the following: (a) χ is quantizable as a Toeplitz quantum map (or Toeplitz Fourier integral operator) if it lifts to a contact transformation χ˜ of (X, α). The quantization is then that of Definition 1.4. (b) χ is quantizable as an automorphism of the full observable algebra if there exists an automorphism α of T ∗ satisfying (1). (c) χ is quantizable as an automorphism of the symbol algebra if there exists an automorphism α of T ∗ /T −∞ satisfying (1). By descending strength, we mean that quantization in the sense above implies quantization in all of the following senses. The automorphisms above are order preserving in the sense that the order of α($A$) is the same as the order of $A$. Henceforth, all automorphisms will be assumed to be order preserving. We now explain the relations between these notions of quantization. We are guided in part by the analogous relations between quantizations of symplectic maps (of cotangent bundles) and automorphisms of the symbol algebra # ∗ /# −∞ of the algebra of pseudodifferential operators, as determined by Duistermaat–Singer in [Duistermaat–Singer (1976)], [Duistermaat–Singer (1975)]. Their main result was that if H 1 (S ∗ M, C) = {0}, then every order-preserving automorphism of # ∗ /# −∞ is either conjugation by an elliptic Fourier integral operator associated to the symplectic map or a transmission (we refer to [Duistermaat–Singer (1976)] for the definition). We prove an analogous theorem for Toeplitz operators and also extend it to the case where the phase space is not simply connected. To state the results, we need some notation. We denote the universal cover of (M, ω) by M˜ and denote the group of deck transformations of the natural cover p : M˜ → M by . We lift all objects on M to M˜ under p. We denote by Tγ the

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˜ We also denote by T ∗ the algebra unitary operator of translation by γ on L2 (M). ˜ of -invariant Toeplitz operators on M. It is important to understand that T∗ is not isomorphic to the algebra of Toeplitz operators on M since there are nontrivial (smoothing) operators which act trivially on automorphic (periodic) functions. In other words, the representation of T∗ on automorphic sections has a kernel, which ˜ we denote by K , and T ∗ (X) ! T∗ (X)/K . Automorphisms which descend to the finite Toeplitz algebras are precisely those which preserve the subalgebra K . For further discussion, we refer to Section 4. Theorem 1.6. With the above notation, we have the following: (0) (Essentially known.) A symplectic map of (M, ω) lifts to a contact transformation of (X, α) and hence defines a Toeplitz quantum map if and only if it preserves holonomies of all closed curves of M. (See Proposition 2.2 of Section 2). (i) Any symplectic map of any compact Kähler manifold (M, ω) is quantizable as an automorphism of the algebra T ∗ /T −∞ of smooth Toeplitz operators over M. (ii) Suppose that H 1 (M, C) = {0}. Then any order-preserving automorphism of T ∗ /T −∞ is given by conjugation with a Toeplitz Fourier integral operator on M associated to a symplectic map χ of (M, α). (The map lifts to a contact transformation of (X, α) by (0)). (iii) Suppose H 1 (M, C) = {0}. Then to each automorphism of T ∗ /T −∞ there corresponds a symplectic map χ of (M, ω) and a Toeplitz Fourier integral operator (Definition 1.5) Uχ on the universal cover M˜ which satisfy Tγ∗ Uχ Tγ = Mγ Uχ , where Mγ is a central operator. The automorphism A → Uχ∗ AUχ is -invariant and defines an order-preserving automorphism of the algebra T∗ which induces α on the -invariant symbol algebra T ∗ /T −∞ . (iv) Let K = ker ρ , where ρ is the representation of T∗ on -automorphic func˜ If α preserves K , then it induces an order-preserving automorphism tions on M. on T ∗ (M) and hence on the finite rank observables OpN (a) on HN . We separate the proof into the cases H 1 (M, C) = {0} in Section 3 and = {0} in Section 4. The latter case is very common in the physics literature on quantum maps. The difference between order-preserving automorphisms of T ∗ and T ∗ /T −∞ is very significant, and only the former automorphisms are quantum maps in the physics sense. For instance, as will be seen in Section 2, Kronecker maps and affine symplectic maps are quantizable as automorphisms of the symbol algebra, but do not lift to contact transformations of X, do not preserve the kernel K and are therefore not automorphisms of T ∗ . Regarding (iv), it is not clear to us whether this operator condition is equivalent to the holonomy-preservation condition in (0). As a corollary, we prove a result which indicates that the physicists’ quantum maps are necessarily Toeplitz quantum maps once they are conjugated to the complex (Bargmann) picture. O Corollary 1.7. If {UN } is a sequence of unitary operators on HN and if UN defines an order-preserving automorphism α of T ∗ /T −∞ , then {UN } must be a Toeplitz H 1 (M, C)


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Fourier integral operator associated to a quantizable symplectic map in the sense of Definition 1.4. As a gauge of our definitions, let us reconsider the Marklof–Rudnick quantizations mentioned above of Kronecker maps, parabolic maps and other “nonquantizable’’ maps [Marklof–Rudnick (2000)]. They define a sequence {UN } of unitary operators on HN satisfying the leading order condition (1), but not to any lower order. Hence conjugation Uχ OpN (a)Uχ∗ of an observable in T ∗ by their quantum map is no longer an observable, i.e., it is not an element of T ∗ . Rather, its Toeplitz symbol only possesses a one term asymptotic expansion and is not a classical symbol. Hence it need not correspond to a quantizable symplectic map. In addition to Theorem 1.6, we discuss a related issue revolving around the quantum maps versus automorphisms distinction: From the viewpoint of quantum chaos, the main interest in the quantum maps Uχ ,N lies in their spectral theory and its relation to the dynamics of χ . This is only well defined when the associated symplectic map is quantizable in the strong sense as a sequence of unitary operators on HN . As stated in the corollary, the symplectic map must then lift to a contact transformation. In the last section Section 6, we point out that even when the symplectic map is quantizable as a unitary operator, it is often the automorphism it induces which is most significant in quantum chaos. That is, much of the spectral theory in quantum chaos concerns the spectrum of the automorphism induced by Uχ ,N rather than the spectrum of Uχ ,N itself.

2 Toeplitz quantization of symplectic maps In this section, we consider the quantization of symplectic maps as Toeplitz Fourier integral operators. In some sense, the material in this section is known, but it seems worthwhile to recall the material and to complete some of the arguments. Suppose that χ : (M, ω) → (M, ω) is a symplectic diffeomorphism. There are several equivalent ways to state the condition that χ is quantizable. The most “geometric’’ one is the following. Definition 2.1. χ is quantizable if χ lifts to a contact transformation χ˜ of (X, α), i.e., a diffeomorphism of X such that χ˜ ∗ α = α. Equivalently, χ lifts to an automorphism of each power LN of the prequantum complex line bundle. It is said to be linearizable in algebraic geometry. Let us consider the obstruction to lifting a symplectic map. We follow in part the discussion in [Guillemin–Sternberg (1977), p. 220]. The key notion is that χ preserves the holonomy map of the connection 1-form α. Recall that the horizontal subbundle H ⊂ T X of the connection is defined by Hx = ker αx = {v ∈ Tx X : αx (v) = 0}. The holonomy map H : → U (1),

H (γ ) = eiθγ

from the free loop space defined by horizontally lifting a loop γ : [0, 1] → M to γ˜ : [0, 1] → X and expressing γ˜ (1) = eiθγ γ˜ (0). We say that χ is holonomy preserving if

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H (χ (γ )) = H (γ )

∀γ ∈ .

If the loop is contained in the domain of a local frame s : U → X, then ∗ H (γ ) = exp 2π i s α .

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γ

If γ = ∂σ , then γ s ∗ α = σ ω. It follows (see [Guillemin–Sternberg (1977)]) that the symplectic map preserves the holonomy around such homologically trivial loops. Hence it is sufficient to consider the map Hχ : H 1 (M, Z) → U (1),

Hχ (γ ) = H (γ )−1 H (χ (γ )) = ei(θγ −θ χ (γ )) . (20)

Proposition 2.2. A symplectic map χ of a symplectic manifold (M, g) lifts to a contact transformation of the associated prequantum S 1 bundle (X, α) if and only if Hχ ≡ 1, the trivial representation. Proof. Suppose that χ lifts to χ˜ : X → X as a contact transformation. Let γ ∈ and let γ˜ be a horizontal lift of γ . Then χ˜ (γ˜ ) is a horizontal lift of χ (γ ). Obviously, γ˜ (1) = eiθγ γ˜ (0) implies χ˜ ◦ γ˜ (1) = eiθγ χ˜ ◦ γ˜ (0), so H = H ◦ χ . Conversely, suppose that Hχ = 1. We then define χ˜ by lifting χ along paths. We fix a basepoint x0 ∈ MX and define χ˜ on the orbit S 1 · x0 by fixing χ˜ (x0 ) to be a chosen basepoint on π −1 (χ (π(x0 )) and then extending by S 1 invariance. We now consider horizontal paths x(t) : [0, 1] → X from x0 . At least one horizontal path exists from x0 to any given point since the curvature is positive (Chow’s theorem). We define χ˜ (x(t)) to be the horizontal lift of χ (π x(t)) to χ˜ (x0 ). To see that this is well defined, we must prove independence of the path. So let x1 (t), x2 (t) be two horizontal paths from x0 to x1 (1). Thus there is trivial holonomy of the loop defined by x1 followed by x2−1 (i.e., the backwards path to x2 ). Now project each path, apply χ , and horizontally lift. This defines a horizontal lift of the loop formed by the projected curves χ ◦ π ◦ xj (t) (j = 1, 2). It has trivial holonomy if χ is holonomy preserving. It follows that the horizontal lifts must agree at t = 1.

As a corollary, we note that for any contact transformation χ of a torus, there exists a unique translation Tα,β so that χ ◦ Tα,β lifts as a contact transformation. Moreover, a contact transformation χ always lifts to a contact transformation if M is simply connected. Hence if we lift χ first to the universal cover M˜ of M, then this further lifts to X˜ as a contact transformation. We verify this in another way, since we will use it in Section 4. ˜ Then there exists a unique (up to Proposition 2.3. Let χ be a symplectic map of M. one scalar) lift χ˜ of χ to X˜ such that π χ˜ = χ π, where π : X˜ → M˜ is the S 1 -fibration. Proof. The fact that χ can be lifted to X˜ is obvious since X˜ ! M˜ × S 1 . The key point is that the map can be lifted as contact transformations. Any lift that commutes with the S 1 action has the form


χ˜ · (z, eiθ ) = (χ (z), eiθ+ϕχ (θ,z) ).

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The contact form on X˜ is the connection 1-form α˜ of the Hermitian line bundle ˜ In local symplectic coordinates (x, ξ ) on M, ˜ it has the form over X. α˜ =

1 (ξ dx − xdξ ) − dθ. 2

˜ and since M˜ is simply connected, Since χ ∗ (xdξ −ξ dx)−(xdξ −ξ dx) is closed on M, ∞ ˜ there exists a function fχ ∈ C (M) such that χ˜ ∗ (xdξ − ξ dx) − (xdξ − ξ dx) = dfχ (x, ξ ). Using the product structure, we have that ϕχ (x, ξ, θ) = fχ (x, ξ ) defines a lift satisfying χ˜ ∗ (α) ˜ = α, ˜ as desired. Regarding uniqueness, the only flexibility in the lift is in the choice of fχ , which is defined up to a constant. The constant can be fixed by requiring that fχ (0, 0) = 0.

There is a weaker condition which has come up in some recent work (see [Marklof–Rudnick (2000)]): Let us say that χ is quantizable at level N if χ lifts to an automorphism of the bundle LN . Often a map is quantizable of level N along an arithmetic progression N = kN0 , k = 1, 2, 3, . . . of powers, although it is not quantizable for all N . In geometric terms, this simply means that χ fails to lift as a contact transformation of X but does lift as a contact transformation of X/ZN , where ZN ⊂ S 1 is the group of N th roots of unity. In everything that follows, the stated results have analogous for this modified version of quantization.

3 Proof of Theorem 1.6 in the case H 1 (M, C) = {0} We first prove that if H 1 (M, C) = {0}, then every automorphism is given by conjugation with a Toeplitz Fourier integral operator. In this case, we may identify maps on M which S 1 -invariant maps on X. We emphasize that we are not considering the most general Toeplitz operators $A$ with A ∈ # ∗ (X) but only the S 1 -invariant operators whose symbols lie in C ∞ (M). The proof is modelled on that of Duistermaat–Singer [Duistermaat–Singer (1976)], but has several new features due to the holomorphic setting. In some respects the proof is simpler, since there are no transmission automorphisms, and there are natural identifications between symbols of different orders. However, in some respects, it is more complicated, and also we must be careful about using contravariant versus covariant symbols. We begin with the following. Lemma 3.1. Suppose that H 1 (M, C) = {0} and that ι is an order-preserving automorphism of T ∞ /T −∞ . Then ι is equal to conjugation by a Toeplitz Fourier integral operator in the sense of Definition 1.4.

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Proof. Since ι is order preserving, it induces automorphisms on the quotients of the filtered algebra T ∗ . We first consider T 0 /T −1 . The map to contravariant symbols defines an identification with C ∞ (M). Thus ι induces an automorphism of C ∞ (M), viewed as an algebra of contravariant symbols under multiplication. The maximal ideal space of C(M) equals M; hence ι induces a map χ on M such that ι(p) = p ◦χ . Precisely as in [Duistermaat–Singer (1976)], one verifies that χ is a smooth diffeomorphism of M. Now consider the quotients T m /T m−1 . They are are simply N m times T 0 /T −1 , so for any m ι(p) = p ◦ χ for p ∈ T m /T m−1 . This step is simpler than in the pseudodifferential case, and as a result certain steps carried out in [Duistermaat–Singer (1976)] are unnecessary here. Now let n = 1, so that T 1 /T 0 is a Lie algebra under commutator bracket. The principal symbol is an isomorphism of the quotient algebra to the Poisson algebra (M, {, }) defined by the symplectic form ω. Since ι is an automorphism of the quotient algebra, we have {a ◦ χ , b ◦ χ } = {a, b} ◦ χ ; hence χ is a symplectic map of (M, ω). This step is also simpler than in [Duistermaat– Singer (1976)], and we see that no transmissions arise as possible automorphisms. By Proposition 2.3, χ lifts to a contact transformation χ˜ of X. 3.0.1 Symbol-preserving automorphisms −1 −1 . It follows Now let A−1 N = $N aTχ $N denote any Toeplitz quantization of χ˜ ∞ −∞ that preserves principal that α(P ) = AN ι(P )A−1 N is an automorphism of T /T contravariant symbols in the sense of Section 1.1.1. We now prove that any such automorphism is given by conjugation with a Toeplitz multiplier of some order s. Thus let j be a principal contravariant symbol-preserving automorphism. Let P ∈ T m . Since j (P ) − P ∈ T m−1 , we get an induced map

βm : C ∞ (M) → C ∞ (M),

βm (a) = j ($N a$N ) − $N a$N .

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Then β = βm is a derivation in two ways: (i) (ii)

β(p · q) = β(p) · q + p · β(q) β({p, q}) = {β(p), q} + {p, β(q)}.

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Now any derivation in the sense of (i) is given by differentiation along a vector field V . Since V commutes with Poisson bracket, it must be a symplectic vector field. Since ω(V , ·) = β is a closed 1-form, there exists a local Hamiltonian H for V . Under our assumption that H 1 (M) = {0}, the Hamiltonian is global, so V = +H for some global H . Thus we have βm (a) = i{a, Hlog bm }

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for some bm ∈ C ∞ (M). Thus j may be represented by j (P ) = B −1 P B for P ∈ T m m ≡ N mS0 , with B = $N eib $N (b = bm ). Because of the natural identification of Sscl scl we find that bm = b is the same for all m. By composing automorphisms, we now have an automorphism j2 such that


j2 ($N aN $N ) − $N aN $N ∈ T m−2 ,

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m aN ∈ Sscl .

We find as above that j2 ($N aN $N )−$N aN $N = β2 (aN ), where β2 is a derivation, hence β2 = N −1 {log b−1 , ·} for some b−1 . Therefore, $N e−iN

−1 b −1

$N j2 (P )$N eiN

−1 b −1

$N − P ∈ T m−2

∀P ∈ T m .

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0 such that Proceeding in this way, we get an element bN ∈ Sscl

$N e−ibN $N j (P )$N eibN $N − P ∈ T −∞

∀P ∈ T m .

This completes the proof of the lemma.

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3.0.2 Conclusion of proof when H 1 (M, C) = {0} Lemma 3 of [Duistermaat–Singer (1976)] is an abstract result which says that automorphisms of Frechet spaces satisfying a certain density condition are always given by conjugation. The density condition is easy to prove, so we omit the proof. The result is the following: Let ι denote an automorphism of T ∗ acting on H ∞ (M). Then ι(P ) = A−1 P A, where A : H ∞ (M) → H ∞ (M) is an invertible, continuous linear map, determined uniquely up to multiplicative constant. Thus i(P ) = A−1 P A for all P ∈ T ∗ , and also, by Lemma 1, there exists an elliptic Toeplitz Fourier integral operator B such that i(P ) ≡ B −1 ◦ P ◦ B for all P ∈ T ∞ /T −∞ . Let E = A ◦ B −1 . Then [E, P ] ∈ T −∞ for all P ∈ T ∞ /T −∞ . In particular, [E, P ] ∈ T −∞ for all P = {$N a$N }, a ∈ C ∞ (M). In place of Lemma 4 of [Duistermaat–Singer (1976)], we use the following. Lemma 3.2. Let E be an operator on H2 such that [E, $a$] ∈ T −∞ for all a ∈ C ∞ (M). Then there exists a constant c such that E = c$+R, where R is a smoothing operator. Proof. It is sufficient to prove the statement for all a supported in a given S 1 -invariant open set U ⊂ X. We can then use a partition of unity to prove the result for all a. We use the notation A ∼U B to mean that A, B are defined on U and their difference is a smoothing operator on U . In a sufficiently small open set U ⊂ X, there exists a Fourier integral operator F : L2 (X) → L2 (Rn ) associated to a contact transformation ϕ such that $ ∼U F $0 F ∗ modulo smoothing operators, where $0 is the model Szegö kernel discussed in [Boutet de Monvel–Sjöstrand (1976)], [Boutet de Monvel–Guillemin (1981)], namely, the orthogonal projection onto the kernel of the annihilation operators Dj = 1i (∂/∂yj + yj |Dt |) on Rn = Rp × Rq . Furthermore, it is proved in [Boutet de Monvel–Sjöstrand (1976)], [Boutet de Monvel–Guillemin (1981)] that there exists a complex Fourier integral operator R0 : L2 (Rq ) → L2 (Rn ) such that R0∗ R0 = I , R0 R0∗ = $0 . Moreover, for any pseudodifferential operator A on X, there exists a

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pseudodifferential operator Q on Rq so that $0 A$0 ∼ R0 QR0∗ . Transporting R0 to X by F , we obtain a complex Fourier integral operator R : L2 (Rq ) → L2 (X) so that RR ∗ ∼U $, R ∗ R ∼ϕ(U ) I and so that $a$ ∼U RQR ∗ . Then [E, $a$] ∼U [E, R ∗ QR] and we may rewrite the condition on E as [E, R ∗ QR] ∈ T −∞ (X)

∀Q ∈ # 0 (Rq ).

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[R ∗ ER, Q] ∈ # −∞ (X)

∀Q ∈ # 0 (Rq ).

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This is equivalent to

We then apply Beals’s characterization of pseuodifferential operators: P ∈ # k (Rm ) if and only if for all {ji , k }, ad(xj1 ) · · · ad(xjr ) ad(Dxk1 ) · · · ad(Dxks )P : H s+r (Rm ) → H s (Rm ) is bounded. Here ad(L)P denotes [L, P ]. It follows first that R ∗ ER ∈ # 0 , and easy symbol calculus shows that the complete symbol of R ∗ ER is constant. Hence R ∗ ER = I + S, where S is a smoothing operator. Applying R on the left and R ∗ on the right concludes the proof.

Remark. It is in the step in Section 3.0.1 that the distinction between symplectic maps of M and contact transformations of X enters. Ultimately it is this step which leads to Corollary 1.7. We also note that the proof above is rather different from that in [Duistermaat–Singer (1976)].

4 H 1 (M, C) = {0} The problems with quantizing symplectic maps on M are all due to the fundamental group π1 (M) or more precisely H1 (M, C). We solve them by passing to the universal ˜ In this section, we relate Toeplitz operators on M and M. ˜ cover M. 4.1 Toeplitz operators on the universal cover Since we are comparing algebras and automorphisms on covers to those on a quotient, we begin with the abstract picture as discussed in [Gromov–Henkin–Shubin (1998)]. We then specialize it to algebras of Toeplitz operators. 4.1.1 Abstract theory Suppose that p : X˜ → X is a covering map of a compact manifold X, and denote its ˜ We would deck transformation group by . We regard as acting on the left of X. ˜ like to compare operators on X and operators on X. To gain perspective, we start ˜ which with the large von Neumann algebra B of all bounded operators on L2 (X) commute with . Later we specialize to the Toeplitz algebra which is our algebra of observables.


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The Schwartz kernel of such an operator satisfies B(γ x, γ y) = B(x, y). If we denote by D a fundamental domain for , then there exists an identification ˜ ! L2 () ⊗ L2 (D) = L2 () ⊗ L2 (X). L2 (X)

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Elements of L2 () ⊗ L2 (X) can be viewed as functions f (γ , x) on × D. The unitary isomorphism is defined by ˜ → fϕ (γ , x) = ϕ(γ · x). ϕ ∈ L2 (X) Note that both left translation Lγ and right translation Rγ by γ act on this space, namely, Lγ f (α, x) = f (γ α, x), Rγ f (α, x) = f (αγ , x). We may regard B as bounded operators commuting with all Lγ . The isomorphism (29) induces an algebra isomorphism B ! R ⊗ B(X),

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where B(X) is the algebra of bounded operators on X and where R is the algebra generated by right translations Rγ on L2 (). ˜ The corresponding algebra So far we have been considering operators on L2 (X). B is much larger than B(X). To make the connection to L2 (X) tighter, we need to ˜ of -periodic functions on X. ˜ The natural Hilbert space consider the space L2 (X) structure is to define f 2 = D |f (x)|2 dV , where dV is a -invariant volume ˜ ! L2 (X). We may regard elements form. We have the obvious isomorphism L2 (X) 2 ˜ as functions f (γ , x) as above which are constant in γ . of L (X) Elements B ∈ B with properly supported kernels, or kernels which decay fast ˜ Indeed, R acts trivially on L2 (X), ˜ so B acts enough off the diagonal, act on L2 (X). by the quotient algebra B /R . We will be working with subalgebras of Toeplitz operators where the action is clearly well defined. Remark. Let us define B as the subalgebra of B of elements which commute with ˜ ! B(X). We may write the (Schwartz) both Rγ and Lγ for all γ . Then we have B (X) kernel of an element of B as B(γ , x, γ , x ). It belongs to B if B(αγ , x, αγ , x ) = B(γ , x, γ , x ), and it belongs to B if addditionally B(γ α, x, α, γ α, x ) = B(γ , x, γ , x ). We have been talking about algebras of bounded operators, but our main interest is in C ∗ -algebras of Toeplitz operators. Everything we have said restricts to these subalgebras once we have defined the appropriate notions. 4.2 Toeplitz operators The positive Hermitian holomorphic line bundle (L, h) → M pulls back under π to ˜ h) ˜ → M. ˜ This induces an inner product on the space H 0 (M, ˜ L˜ N ) of entire one (L,

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˜ L˜ N ) the space of L2 holomorphic holomorphic sections of L˜ N . We denote by H2 (M, sections relative to this inner product. As in the quotient, there exists an associated S 1 bundle X˜ with a contact (connection) form α˜ such that X˜ → M˜ ↓ ↓ X→M commutes. The vertical arrows are covering maps and the horizontal ones are S 1 ˜ It is isomorphic bundles. We denote the deck transformation group of X˜ → X by . to , so when no confusion is possible we drop the˜. Since all objects are lifted from quotients, it is clear that ˜ acts by contact transformations of α. ˜ Let us the denote operator of translation by γ on M˜ by Lγ . ˜ the Hardy space of L2 CR functions on X. ˜ They are boundary We denote by H2 (X) values of holomorphic functions in the strongly pseudoconvex complex manifold D˜ ∗ = {(z, v) ∈ L˜ ∗ : hz (v) < 1},

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˜ The group ˜ acts on D˜ ∗ ⊂ L˜ ∗ with quotient the compact disc bundle which are L2 (X). ∗ ∗ D ⊂ L → M. In this setting it is known (see [Gromov–Henkin–Shubin (1998), Theorem 0.2]) that ˜ = ∞. dim H2 (X) Due to the S 1 symmetry, holomorphic functions on D˜ ∗ are easily related to CR ˜ We denote by holomorphic functions on X. ˜ → H2 (X) ˜ ˜ : L2 (X) $

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the Szegö (orthogonal) projection. Under the S 1 action, we have ˜ = H2 (X)

∞ D

2 ˜ HN (X),

˜ = $

N =1

∞ D

˜ N. $

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N =1

2 (X) ˜ ! H2 (M, ˜ L˜ N ). We refer to [Gromov–Henkin–Shubin (1998), As on X, we have HN example (2), p. 559] for the proof that L˜ → M˜ has many holomorphic sections. ˜ More important are periodic funcSo far we have discussed L2 functions on X. tions. We endow them with a Hilbert space structure by setting + ˜ = {f ∈ L2 (X) ˜ : Lγ f = f }, L2 (X) loc (34) 2 2 ˜ ˜ H (X) = {f ∈ L (X), ∂ b f = 0},

with the inner product , obtained by integrating over a fundamental domain D 2 (X) ˜ for the S 1 action for . Both are direct sums of weight spaces L2,N , resp. H,N 2 ˜ There exists a Hilbert space isomorphism L : H (X) ˜ = H2 (X), namely, by on X. ∗ lifting Lϕ = p ϕ under the covering map. The adjoint of L is given by L∗ f = p∗ (f 1D ). We thus have


˜ → H2 (X). ˜ LL∗ = Id : H2 (X) 2 (X) ˜ H,N

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2 (X) ˜ HN

We observe that the spaces and are completely unrelated and have different dimensions. The former is canonically isomorphic to HN (X). We now consider Toeplitz algebras. Since X˜ is noncompact and infinite volume in general, we must take care that Toeplitz operators are well defined and form an algebra. As for pseudodifferential operators on infinite volume spaces, we define ˜ as the space of operators of the form $A ˜ is the space of ˜ $, ˜ where A ∈ # s 1 (X) T s (X) S 1 properly supported pseudodifferential operators commuting with S . We also define ˜ $ ˜ with A having a smooth properly supported kernel. T −∞ as the space of such $A ˜ off the diagonal (see (36)), the operators $A ˜ $ ˜ Due to the exponential decay of $ have exponentially decaying kernels (relative to the -invariant volume form) and have well-defined compositions. We then distinguish the automorphic Toeplitz operators ˜ = {$A ˜ : L∗γ $A ˜ $L ˜ γ = $A ˜ $ ˜ ∈ T ∗ (X) ˜ $}. ˜ T∗ (X) ˜ = 0 or, equivalently, $(γ ˜ x, γ y) = $(x, ˜ We note that [Lγ , $] y). So the operative condition is that A ∈ #S 1 , , the space of pseudodifferential operators commuting ˜ with . The associated symbols aN (z, z¯ ) are exactly the -invariant symbols on M. We note the following. ˜ on H2 preserving Proposition 4.1. There exists a representation ρ of T∗ (X) 2 each H,N . Proof. Since Lγ $A$f = $A$f whenever Lγ f = f , the only issue is whether Af is well defined for f ∈ H . However, A is a polyhomogeneous sum of aj N −j ,

where aj is a periodic function, so the action is certainly defined. Let us denote by K = ker ρ . We further denote by ρ,N the associated repre2 , and put K = ker ρ sentation on H,N ,N . ˜ Proposition 4.2. K ⊂ T −∞ (X). ˜ annihilates H2 (X) ˜ ! H2 (X). This means that Proof. Assume that $A$ ∈ T∗ (X) ˜ In particular it implies that the “Berezin symbol’’ Af, gD = 0 for all f, g ∈ H2 (X). ˜ N aN $ ˜ N (z, z) = 0. However, asymptotically, N −m $ ˜ N aN $ ˜ N (z, z) ∼ a0 (z) for $ a zeroth-order Toeplitz operator. One sees by induction on the terms in (10) that A ∼ 0.

It could happen that K = 0, unlike the analogous representation on H2 (X) which defines Toeplitz operators. For each N there could exist aN ∈ C ∞ (M) with 2 (X) ˜ ! H2 (X) aN L2 = 1 which is orthogonal to the finite-dimensional space H,N N 2 (X). ˜ Then T = $ ˜ N aN $ ˜ N ∈ K,N . but which is not orthogonal to HN ˜ to T ∗ (X). In preparation, we relate the Szegö kernels on We now relate T∗ (X) ˜ First, we consider a fixed N . The following is proved in [Shiffman–Zelditch]. X, X.

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Proposition 4.3. The degree N Szegö kernels of X, X˜ are related by ˜ N (γ · x, y). $ $N (x, y) = γ ∈ 2 . The same formula defines the Szegö projector L2,N → H,N

A key point is to use the estimate √ ˜ N d(x,y)

˜ N (x, y)| ≤ Ce− |$

,

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˜ y) is the Riemannian distance with respect to the Kähler metric ω˜ to show where d(x, ˜ N acts on that the sum converges for sufficiently large N . The estimates show that $ ˜ Since L2 (X) ˜ ∩ C(X) ˜ ⊂ L∞ (X), ˜ $ ˜ and we have ˜ N acts on H 2 (X), L∞ (X). ˜ N (x, y)sN (y)dV (y) = ˜ N (x, γ y)sN (y)dV (y). ˜ N sN (x) = $ $ $ X˜

D γ ∈

˜ ˜ N = sN for sN ∈ H 2 (X). To complete the proof, one has to prove that $s Now we consider the full Szegö kernel. ˜ N L for each N as operators from L2 (X) to H2 . Corollary 4.4. We have L$N = $ N ,N 2 2 ˜ ˜ : L (X) → H (X). Hence L$ = $L ˜ The identity (30) for the larger algebra of bounded operators suggests that T∗ (X) should be a larger algebra than T ∗ (X). However, this is not the case. ˜ ˜ Proposition 4.5. L induces an algebra isomorphism T ∗ (X) ! T (X)/K (X). Proof. It follows from Proposition 4.1 and Corollary 4.4 that ˜ ˜ : L2 (X) → H2 (X) ˜ ∗ a $L L$a$ = $p ˜ : L2 (X) → H2 (X). ˜ ∗ a $L ⇐⇒ $a$ = L∗ $p

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Equality on the designated spaces is equivalent to equality in the algebras. Further, the equality LL∗ = I : H2 → H2 implies that the linear isomorphism is an algebra isomorphism.

˜ is so small. We recall that one obtains T ∗ (X) It may seem surprising that T (X) 2 ˜ on H (X). ˜ When dealing with all bounded operators, the by representing T (X) kernel is very large (R ) and it is also large if we fix N and consider the associated Toeplitz algebra. But the kernal is trivial if we consider the full Toeplitz algebra. We also have the following. ˜ Corollary 4.6. L induces algebra isomorphisms TN (X) ! T,N (X)/K ,N . ˜ The concrete Now let us relate such automorphisms to automorphisms on X. identification with T (X) is by (37). We have the following. Proposition 4.7. There is a natural identification of •

˜ automorphisms α on T ∗ (X) with automorphisms α˜ on T∗ (X)/K ;


•

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−∞ ˜ automorphisms α on T ∗ (X)/T −∞ (X) with automorphisms α˜ on T∗ (X)/T .

Proof. The first statement is clear since the algebras are isomorphic.An automorphism of T∗ descends to T ∗ if and only if it preserves K . Concretely, we wish to set ˜ ∗ a $)L. ˜ α($a$) = L∗ α( ˜ $p

(38)

The inner operator must be determined by the left side for this to be well defined. We have ˜ ∗a$ ˜ ≡ L$a$L∗ mod K . $p (39) The same equivalence is true modulo the larger subalgebra T−∞ . Since T−∞ /K = T −∞ (X), the second statement is correct.

4.3 Completion of the proof of Theorem 1.6 We now prove statements (iii)–(iv) of the theorem. The following gives an upper bound on existence of semiclassical automorphisms. Lemma 4.8. Suppose that α is an order-preserving automorphism of T ∗ (X)/T −∞ . ˜ Let α˜ denote the corresponding automorphisms of T∗ (X)/K . Then there exists a canonical transformation χ of (M, ω) and a unitary Toeplitz quantum map U˜ χ on ˜ such that H 2 (X) α(P ˜ ) = U˜ χ∗ P U˜ χ and such that

˜ ˜ L−1 γ U χ L γ = Mγ U χ ,

˜ where Mγ commutes with T∗ (M). Proof. By Lemma 3.1, we know that α˜ is given by conjugation by a Toeplitz quantum map U˜ χ . We may define Mγ by the formula above since U˜ χ is invertible. We then determine its properties. We have −1 ˜ ˜ −1 ˜ −1 ˜ L−1 γ U χ L γ P L γ Uχ L γ = U χ P U χ

˜ ∀P ∈ T∗ (M).

Hence Mγ−1 U˜ χ−1 P U˜ χ Mγ = U˜ χ−1 P U˜ χ ⇐⇒ Mγ−1 P Mγ = P It follows that Mγ is central. This proves (iii) of Theorem 1.6.

˜ ∀P ∈ T∗ (M).

The lower bound is given as follows. Lemma 4.9. Suppose that χ is a symplectic map of (M, ω). Then it lifts to a con˜ α). tact transformation χ˜ of (X, ˜ The associated quantum map Uχ˜ on X˜ defines (by ˜ which descends to an conjugation) an order-preserving automorphism α˜ of T (X) automorphism of T ∗ (X)/T −∞ . If α˜ preserves K , then it defines an automorphism of all of T ∗ (X). Proof. χ automatically lifts to M˜ as a symplectic map commuting with the action of . By Proposition 2.3 it lifts to X˜ as a contact transformation. We then define a unitary quantum map by

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˜ N σ Tχ˜ $ ˜ N, U˜ N χ˜ = $ ˜ See where σ is a function on M˜ which makes the operator unitary on H2 (X). [Zelditch (1997)] for background. ˜ When χ A crucial issue now is the commutation relations between U˜ N χ˜ and . ˜ lifts to X, i.e., is quantizable, then χ˜ commutes with . In this case, χ is quantizable as a quantum map and there was no need to lift it to X˜ to quantize it as an automorphism. Assume, however, that χ does not lift to X and consider the commutation relations ˜ The commutator of the translation by χ˜ with left translations by elements of . −1 −1 ˜ ˜ χ˜ γ˜ χ˜ γ˜ covers the identity map of M since the lift of χ to M commutes with . ˜ It follows that Furthermore, it commutes with the S 1 action on X. χ˜ γ˜ χ˜ −1 γ˜ −1 = Teiθγ ,χ ,

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where the right side is translation by the element eiθγ ,χ . The angle θγ ,χ is a priori a ˜ However, the left side is a contact transformation covering the identity function on M. and therefore dθ = dθ + dθγ ,χ , i.e., θγ ,χ is a constant. After quantizing, the same commutator identity holds for the operators. Therefore the operators Mγ are central. It follows that the automorphism α(P ˜ ) = U˜ χ∗ P U˜ χ satisfies

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˜ ˜ N p ∗ aN $ ˜ N ) ∈ T∗ (X). α˜ N ($

It therefore descends to T ∗ (X)/T −∞ (X) by (38), i.e., as ˜ N p ∗ aN $ ˜ N ) = L∗ U˜ χ∗ $ ˜ N p ∗ aN $ ˜ N )U˜ χ L. α˜ N ($ Unitarity of L then implies that α is also an automorphism. If the automorphism preserves K , then it also descends to T ∗ (X).

An obvious question is whether the condition that the automorphism preserve K is equivalent to the quantization condition that χ lift to X. Clearly, quantizability in the sense of Definition 1.5 implies preservation of K , since the quantum map Uχ ,N is well defined on the spaces HN . The converse is not obvious, since we only know a priori that the automorphism induces automorphisms αN of the finite rank observables OpN (aN ) for fixed N . Abstractly, such automorphisms must be given by conjugations by unitary operators on HN , but it is not clear that these unitary operators are Toeplitz quantum maps in the sense of Definition 1.5. We end the section with the following proof. Proof of Corollary 1.7. This follows immediately from (ii) if H 1 (M, C) = {0}. If H 1 (M, C) = {0}, then by Theorem 1.6(iii) there exists a symplectic map χ of M and a Toeplitz Fourier integral operator V˜χ on M˜ and a central operator Mγ such that Tγ∗ V˜χ Tγ = Mγ V˜χ , and such that α is induced by conjugation by V˜ . But by definition, α is also given by conjugation by U . Now the Schwarz kernel of U , hence U , lifts to


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˜ By assumption, U˜ AU˜ ∗ has the same complete symbol a -invariant kernel U˜ on M. ∗ ˜ ˜ as V AV for any Toeplitz operator A on M, lifted to T . By Lemma 3.2, it follows that U˜ = V˜ + R, where R is a smoothing Toeplitz operator. It follows that Mγ = 1 (hence θγ ,χ = 1 for all γ ), and therefore the symplectic map χ˜ underlying V˜ , when ˜ is invariant under the deck transformation group ˜ of X˜ → X. lifted to X,

5 Quantization of torus maps To clarify the issues involved, we consider some standard examples on the symplectic 2m-torus T2m = Cm /Z2nm . Since H1 (T2m , C) = C2m , there will exist symplectic maps which cannot be quantized in the sense of Definitions 1.4 and 1.5(a) as quantum maps, though they can and will be quantized as automorphisms. In fact, the distinction can already be illustrated with the simplest maps: • •

Kronecker translations Tθ (x) = x + θ (x, θ ∈ T2m ); symplectic automorphisms A ∈ Sp(2m, Z).

We begin by describing the line bundle on the torus and its universal cover. We follow [Zelditch (1997)], [Bleher–Shiffman–Zelditch (2001)] and refer there for further discussion. The quotient setting is L → T2n , where L is the bundle with curvature j dzj ∧ d z¯ j . Sections of LN are theta-functions of level N . On the universal cover, we have the pulled back bundle LH = C × Cm → Cm . Its associated principal S 1 bundle m . We recall that it is the quotient Cm ×S 1 → Cm is the reduced Heisenberg group Hred under the subgroup (0, Z) in the center of the simply connected Heisenberg group Hm = Cm × R with group law 1 (ζ, t) · (η, s) = (ζ + η, t + s + 4(ζ · η)). ¯ 2 The identity element is (0, 0) and (ζ, t)−1 = (−ζ, −t). The reduced Heisenberg m = Hm /{(0, k) : k ∈ Z} = Cm × S 1 with group law group is thus Hred 1

¯ (ζ, e2π it ) · (η, e2π is ) = (ζ + η, e2π i[t+s+ 2 4(ζ ·η)] ). m with the left-invariant connection form We now equip Hred

αL =

1 dt (ξq dxq − xq dξq ) − 2 q 2π

(ζ = x + iξ ),

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whose curvature equals the symplectic form ω = q dxq ∧ dξq . The kernel of α L is the distribution of horizontal planes. To define the Szegö kernel, we further need to split the complexified horizontal spaces into their holomorphic and antiholomorphic parts. The left-invariant (CR-)holomorphic (respectively, antiholomorphic) vector m are the horizontal lifts of the vector fields ∂ , fields ZqL (respectively, Z¯ qL ) on Hred ∂zq

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respectively,

∂ ∂ z¯ q

m ) of CR with respect to α L . We then define the Hardy space H2 (Hred

m ) satisfying the left-invariant holomorphic functions to be the functions in L2 (Hred m . For N = 1, 2, . . . , we L ¯ Cauchy–Riemann equations Zq f = 0 (1 ≤ q ≤ m) on Hred m 2 2 further define HN ⊂ H (Hred ) as the (infinite-dimensional) Hilbert space of squareintegrable CR functions f such that f ◦ rθ = eiN θ f as before. The representation H12 is irreducible and may be identified with the Bargmann–Fock space of entire 2 holomorphic functions on Cn which are square integrable relative to e−|z| . The H 2 Szegö kernel $N (x, y) is the orthogonal projection to HN . It is given by

$H N (x, y) =

1 m iN (t−s) N (ζ ·η− ¯ 12 |ζ |2 − 12 |η|2 ) N e e , m π

x = (ζ, t),

y = (η, s).

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We note that it satisfies the estimates in (36). In this model example, Proposition 4.3 was proved in [Zelditch (1997)]. Finally, we describe the circle bundle X in the quotient setting. The lattice Z2m m of Hm under the homomorphism may be embedded as a subgroup HZ R ι(m, n) = (m, n, eiπ m·n ).

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m . To clarify the role of the factors of 1 , we show that We will denote the image by HZ 2 m HZ is indeed a subgroup:

(m, n, eiπm·n ) · (m , n , eiπ m ·n )

= (m + m , n + n , eiπ(m·n+m ·n +mn −m n) ) = (m + m , n + n , eiπ(m·n+m ·n +mn +m n) )

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= (m + m , n + n , eiπ((m+m )·(n+n )) ). m . The leftWe then put X = HZm \H n mR , i.e., X is the left quotient of HRm by HZ L invariant contact form α descends to X as a contact form and a connection form for the principal S 1 bundle X → Cm /Z2m .

5.1 Kronecker translations We first show that irrational Kronecker translations T(a,b) f (x, ξ ) = f (x + a, ξ + b)

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are nonquantizable as Toeplitz quantum maps. Proposition 5.1. T(a,b) fails to be quantizable for all (a, b) ∈ R2n /Z2n . T(a,b) is quantizable at level N iff N a, N b ∈ Z2n . Proof. By Proposition 2.2, the map lifts if and only if translations preserve holonomy of homologically nontrivial loops. The loops on T2m that we need to consider are


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given in local coordinates by γm,n (t) = (tm, tn). Horizontal lifts to X are given by γ˜m,n (t) = (tm, tn, 1). At t = 1 we obtain (m, n, 1) ∼ (0, 0, eiπ m·n ). Hence the holonomy of the path γm,n equals eiπ m·n . Now translate the loop γ(m,n) by (a, b) to obtain the loop γ1 (t) = (tm+a, tn+b). A horizontal lift to X is given by γ˜1 (t) = (tm + a, tn + b, eπ i(b·m−a·n)t ). It is the projection to X of the left translate by (a, b, 0) of the original horizontal path. At t = 1 the endpoint is (m + a, n + b, eπ i(b·m−a·n) ) = (a, b, eiπ[m·n+2(b·m−a·n)] ). Hence the holonomy changed by e2π i(b·m−a·n) . The holonomy is preserved iff b · m − a · n ∈ Z for all (m, n) ∈ Z2m iff (a, b) ∈ Z2m . Lifting to level N means changing the holonomy to e2π iN θγ . So the condition to lift becomes (a, b) ∈ N1 Z2 .

Remark. The nonquantizability of T(a,b) is due to the left–right invariance of various objects. T(a,b) only lifts to HZ \HR as right translation by (a, b, 0). But right translation by an element of HR does not preserve the left invariant contact form. Equivalently, T(a,b) only lifts to a contact transformation of HR if it lifts to left translation by (a, b, 0). But then the lift does not descend to HZ \HR . 5.1.1 Kronecker translations as automorphisms It is easy to see that Kronecker translations define automorphisms of the revelant algebras. We lift T(a,b) to HRn as the contact transformation of left multiplication T(a,b) (x, ξ, e2π it ) := (x + a, ξ + b, e2π it eπ i(aξ −bx) ).

Although the map T(a,b) does not descend to the quotient as a map, we claim the following. Proposition 5.2. Kronecker maps T(a,b) have the following properties: (i) T(a,b) defines an automorphism of T∗ . (ii) T(a,b) defines an automorphism of T ∞ (X)/T −∞ (X) by αa,b;N (OpN (a)) = OpN (a ◦ T(a,b) ). (iii) However, α(a,b) does not preserve K and does not define an automorphism of T ∞ (X). Proof. (i) Left translation by (a, b) defines an automorphism of T∗ because, by (43), the Szegö kernel commutes with left translations, i.e., H $H N (α · x, α · y) = $N (x, y) ∀α.

(47)

Indeed, it is the kernel of a convolution operator. T , where γ ∈ = Z2m . An easy computa(ii) Consider the conjugates Tγ−1 Ta,b γ tion shows that

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S. Zelditch Tγ−1 Ta,b Tγ f (x, ξ, t) = Mγ Ta,b f (x),

where Mγ f (x, ξ, t) = f (x, ξ, t + ω(γ , (a, b)). ˜ Nσ$ ˜ N with We need to show that Mγ commutes with every Toeplitz operator $ symbol lifted from Cm /Z2m . Since the symbol is invariant under the central circle, it ˜ N ] = 0. But this follows as long as $ ˜ N (z · x, z · y) = is sufficient to show that [Mγ , $ it 1 ˜ $N (x, y) for any z = e ∈ S , the center of the Heisenberg group. But this follows because ˜ N (z · x, z · y) = |z|2N $ ˜ N (x, y). ˜ N (x, y) = $ $ ˜ N , the automorphism descends to the Since left translation commutes with $ quotient as

∗ ˜ ˜ N )Tα,β ($N p ∗ aN $ L αN ($N aN $N ) = L∗ Tα,β ˜ N (Ta,b ˜ N L. = L∗ $ p ∗ aN )$

This is the stated formula. (iii) A Kronecker automorphisms α(a,b) can only preserve K,N if $N a$N = 0 implies $N (a ◦ Ta,b )$N = 0. But if this were the case, the elements $N eik,x $N would be distinct eigenoperators with eigenvalues eik,(a,b) . This contradicts the finite dimensionality of the algebra for fixed N .

5.2 Quantum cat maps We now show, in a similar way, that symplectic linear maps of T2 always define quantum automorphisms even though they do not always define quantum maps. We write ab g= ∈ SL(2, Z), c d and define g(x, ξ ) = (ax +bξ, cx +dξ ) on the torus. It lifts to the reduced Heisenberg group by g(x, ξ, t) = (g(x, ξ ), t). Proposition 5.3. Tg is quantizable iff a · c, b · d ∈ 2Z. Proof. We go through the same calculation as for Kronecker translations. This time, the horizontal lift of the transformed loop is (t (a · m + b · n), t (c · m + d · n), 1). At t = 1, the endpoint is ((a · m + b · n), (c · m + d · n), 1) = (0, 0, eiπ(a·m+b·n)·(c·m+d·n) ). Since the holonomy of the original path was eiπ m·n , the change in holonomy equals eiπ(m·n−(a·m+b·n)(c·m+d·n)) = 1 ⇐⇒ ac, bd ∈ 2Z. Here we use that ad + bc ≡ 1(mod 2Z).


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5.2.1 Linear maps as automorphisms It is known that quantizable linear maps (cat maps) on the quotient define quantum maps with exact Egorov theorems (see, e.g., [Zelditch (1997)]). We now show that nonquantizable maps as well-defined automorphisms by the exact Egorov formula. Proposition 5.4. Tg defines an automorphism of T ∞ (X)/T −∞ (X) by αg;N (OpN (a)) = OpN (a ◦ Tg ). Proof. Consider the conjugates Tγ−1 Tg Tγ , where γ ∈ . We have Tγ−1 Tg Tγ f (x, ξ, t) = Mγ Tg f (x), where Mγ f (x, ξ, t) = f ((x, ξ ) + (I − g)γ , t + ω(γ , z) − ω(γ , g(z + γ )). Mγ is the composition of translation T(I −g)γ with a central translation. Since (I −g)γ is in the lattice, translation by this element commutes with left invariant operators. ˜ . Thus Mγ ∈ T∗ (X) Thus the automorphism descends to the quotient as ˜ N p ∗ aN $ ˜ N )Tg L αN ($N aN $N ) = L∗ Tg∗ ($ ˜ N L. ˜ N (Tg p ∗ aN )$ = L∗ $

6 Spectra of automorphisms In this article, our interest lies in the automorphisms defined by symplectic maps. But most of the interest in quantizations of quantizable symplectic maps, at least in the physics literature, is in their spectral theory as unitary operators Uχ ,N on the finite-dimensional Hilbert spaces HN (X). In this section, we point out how the most important aspects of this spectral theory of U pertain only to the spectrum of the associated automorphism U AU ∗ . The main point is that the reformulation suggests generalizations to other kinds of automorphisms. We also tie together the automorphisms of Toeplitz algebras on the torus with the well-known ones on the rotation algebra. 6.1 Spectra of automorphisms of Hilbert–Schmidt algebras We let H denote a Hilbert space, and denote by HS the algebra of Hilbert–Schmidt operators on H, i.e., the operators for which the inner product A, B := Tr AB ∗ is finite. We let ∗ denote the adjoint on H; no confusion with the ∗ for the star product should arise. A finite-dimensional algebra of Hilbert–Schmidt operators is of course a full matrix algebra, and its automorphisms are given by conjugation by unitary operators. Suppose that α is an automorphism of HS.

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Definition 6.1. We say that an automorphism α of HS is • • • •

a ∗-automorphism if α(A∗ ) = α(A)∗ ; unitary if α(A), α(B) = A, B; a conjugation if there exists a unitary operator U : H → H s.t. α(A) = U AU ∗ ; tracial if Tr α(A) = Tr A for all A of trace class.

We will consider the eigenvalues and “eigenoperators’’ of a unitary ∗-automorphism on HS: α(A) = eiθ A. If α is a unitary automorphism, then (as a unitary operator) it possesses an orthornormal basis of eigenoperators {Aj }. The following is elementary from the definitions. Proposition 6.2. We have the following: (i) A tracial ∗-automorphism is unitary. (ii) The composition of any two eigenoperators is a (possibly zero) eigenoperator. (iii) If Aj is an eigenoperator, then A∗j Aj is an invariant operator, i.e., α(A∗j Aj ) = A∗j Aj . Proof. (i) This is immediate from the fact that α(A), α(B) = Tr α(A)α(B)∗ = Tr α(AB ∗ ) = Tr AB ∗ = A, B. (ii)–(iii) These statements follow from the equations α(Aj Ak ) = α(Aj )α(Ak ) = ei(θj +θk ) Aj Ak , and α(A∗j ) = [α(Aj )]∗ = e−iθj α(A∗j ).

In the case α(A) = U ∗ AU we note that the eigenoperators of the automorphism are given by ∗ ∗ α(ϕN,j ⊗ ϕN,k ) = ei(θN,j −θN,k ) (ϕN,j ⊗ ϕN,k ), (48) where {(ϕN,j , eiθN,j )} are the spectral data of U . 6.2 Spectral problems of quantum chaos The main problems on quantum maps pertain to the spacings between eigenvalues (the pair correlation problem) and the asymptotics of matrix elements relative to eigenfunctions of the operators. 6.2.1 Pair correlation problem Let us recall that the pair correlation function ρ2N (PCF) of a quantum map {UN } with Planck constant 1/N is the function on R defined by ∞ ˆ f (x)dρ2N (x) = f | Tr UN |2 . N R =0

Its limit as N → ∞, when one exists, is the PCF of the quantum map. Clearly,


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knowledge of dρ2N is equivalent to knowledge of its form factor | Tr UN |2 . We observe that the form factor depends only on the automorphism below. Proposition 6.3. The form factor of a conjugation automorphism {αN } is given by = αN Aj , Aj , Tr αN j

where {Aj } is an orthonormal basis for HS N . = U ⊗ U − on HS , and we have Indeed, if α(A)N = UN∗ AUN , then αN N N N − 2 Tr HS N UN ⊗ UN = | Tr HN UN | . Hence the pair correlation problem makes sense for all unitary automorphisms αN .

Problem. Given any unitary automorphism αN , determine N → ∞, where αN (j ) = eiϑN,j j

1 dN

dN2

j =1 δ(N (ϑN,j )) as

(49)

is the eigenvalue problem for the automorphism. 6.2.2 Problems of quantum ergodicity/mixing We observe that these too can be formulated for any sequence of automorphisms. We ∗ as the rewrite the asymptotics of matrix elements AϕN,j , ϕN,k = Tr AϕN,j ⊗ ϕN,k ∗ inner products A, j k . We observe that the eigenfunctions k,k = ϕN,k ⊗ ϕN,k always have eigenvalue 1, i.e., they are invariant states of the automorphism. It is simple to check that the proof of quantum ergodicity for quantizations of ergodic quantizable symplectic maps χ (see [Zelditch (1997)]) uses only the automorphism involved. It states that if a symplectic map χ is ergodic and quantizable, then the invariant states of the corresponding automorphism of the Toeplitz algebra are asymptotic to the traces τN (A) = dim1HM Tr A|HN . It might be interesting to find generalizations of this result to other kinds of automorphisms. 6.3 Spectral theory of model automorphisms We now point out that the automorphisms induced by model quantum maps on the torus are the same as the well-known automorphism of the finite-dimensional rotation algebras. 6.3.1 The rotation algebra modulo N We denote by GN the finite Heisenberg group of order N 2 , generated by two elements U, V satisfying U2 U1 = e2π i/N U1 U2 ,

U1N = U2N = I,

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and its group algebra by RN . GN has a unique irreducible unitary representation ρN on CN given as follows: If we regard CN = L2 (Z/NZ), then ρN (U1 )ψ(Q) = e

2π iQ N

ψ(Q),

ρN (U2 )ψ(Q) = ψ(Q + 1).

Recall that the rotation algebra or noncommutative torus Aθ is the (pre-)C ∗ -algebra generated by unitaries U1 , U2 satisfying the Weyl commutation relation U2 U1 = e2π iα U1 U2 . When α = 1/N, Aθ has a large center generated by U1N , U2N . RN is obtained from Aθ by viewing central elements as scalars. 6.3.2 Toeplitz algebra and rotation algebra We identify the rotation algebra with θ = 2π N to the algebra of Toeplitz operators $N a$N on the torus. As verified by S. Nonnenmacher [Nonnenmacher (2003)], the elements 2 2 U1 = eπ N $N eiθ1 $N , U2 = eπ N $N eiθ2 $N (50) satisfy UjN = I . Here (eiθ1 , eiθ2 ) are the standard coordinates on the torus. Hence any quantum map on the torus defines an automorphism of RN . Thus we can identify the automorphisms αg,N quantizing ab g= c d with the well-known automorphisms of RN defined by U1 → U1a U2b , U2 → U1c U2d (see, e.g., [Narnhofer (1997)]). We can also see easily from this point of view that Kronecker maps Tu,v cannot in general be quantized as automorphisms. Namely, the quantization on R2 translates the symbol, so it would descend to U1 → eiu U1 , U2 → eiv U2 . To be well defined, one needs eiu , eiv to be N th roots of unity, which of course they are not in the irrational case.

7 Appendix The key elements of the Toeplitz algebra and its automorphisms are the ∗ product (13) and the Egorov formula (1). The purpose of this appendix is to direct the reader’s attention to the existence of routine calculations of the complete symbols of compositions aN ∗N bN of symbols and of conjugations UN OpN (a)UN∗ of observables by Toeplitz quantum maps. The method is to use the Boutet de Monvel– Sjöstrand parametrix for the Szegö kernel [Boutet de Monvel–Sjöstrand (1976)] as in [Zelditch (1998)]. Since the original version of this paper was written, several papers [Karabegov–Schlichenmaier (2001)], [Schlichenmaier (1999)], [Schlichenmaier (1998)], [Schlichenmaier (1999b)], [Shiffman–Tate–Zelditch (2003)] have also used this method to describe Toeplitz ∗ product on symbols, so we only briefly mention how to go about calculating asymptotic expansions.


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Proposition 7.1. Let (M, ω) be a compact Kähler manifold. Then the ∗ product defines an algebra structure on classical symbols. There exists an asymptotic expansion fˆ1 ∗ fˆ2 (z, z¯ ) ∼

∞

N −k Bk (f1 , f2 ),

k=0

where B0 (a, b) = f1 · f2 , B1 (f1 , f2 ) = 12 {f1 , f2 } and where Bk is a bidifferential operator of C ∞ (M) × C ∞ (M) → C ∞ (M). Proof. Using the Boutet de Monvel-Sjostrand parametrix as in [Zelditch (1997)], [Shiffman–Tate–Zelditch (2003)], one can obtain a complete asymptotic expansion of the covariant symbol $N a$N b$N (z, z¯ ). One writes out $N (z, w) as an oscillatory integral and applies complex stationary phase. For calculations of this kind, we refer to [Shiffman–Tate–Zelditch (2003)]. To obtain a ∗N b, we invert the Berezin transform IN on symbols, as described in [Reshetikhin–Takhtajan (1999)] and elsewhere. It is invertible on formal power series, and the same inverse is well defined on symbol expansions. Thus a ∗N b ∼ IN−1 $N a$N b$N (z, z¯ ). This produces the symbol expansion claimed in the proposition.

Proposition 7.2. Let Uχ ,N be a Toeplitz quantum map as in Definition 1.5. Then for any observable $N aN $N = OpN (aN ), the contravariant symbol aχ of Uχ∗,N OpN (aN )Uχ ,N possesses a complete asymptotic expansion aχ (z) ∼

∞

N −k Vk (a ◦ χ ),

k=0

where V0 (a) = a, and where Vk is a differential operator of order at most 2k. Proof. The expansion is obtained from the covariant symbol Uχ∗,N OpN (aN )Uχ ,N (z, z¯ ) by inverting the Berezin transform. The asymptotics of the covariant symbol follow by applying stationary phase to the oscillatory integral formula for Uχ∗,N OpN (aN )Uχ ,N .

Acknowledgments The author would like to thank S. de Bievre, Z. Rudnick, and particularly S. Nonnenmacher for helpful discussions on this paper during the program on Semiclassical Methods at MSRI in Spring, 2003. The author would also like to thank the Clay Mathematics Institute for partial support during this period.

References [Berezin (1972)] F. A. Berezin, Covariant and Contravariant symbols of operators, Math. USSR Izvest., 6 (1972), 1117–1151.

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[Berezin (1974)] F. A. Berezin, Quantization, Math. USSR Izvest., 8 (1974), 1109–1165. [Bleher–Shiffman–Zelditch (2001)] P. Bleher, B. Shiffman, and S. Zelditch, Universality and scaling of zeros on symplectic manifolds, in Random Matrix Models and Their Applications, Mathematical Sciences Research Institute Publications, Vol. 40, Cambridge University Press, Cambridge, UK, 2001, 31–69. [Boutet de Monvel 1 (1999)] L. Boutet de Monvel, Star-produits et star-algèbres holomorphes, in G. Dito and D. Sternheimer, eds., Conférence Moshé Flato 1999: Quantization, Deformations, and Symmetries, Vol. I, 1999, Mathematical Physics Studies, Vol. 21, Kluwer Academic Publishers, Dordrecht, The Netherlands, 2000, 109–120. [Boutet de Monvel 2 (1998)] L. Boutet de Monvel, Star produits holomorphes, in Séminaire: Equations aux Dérivées Partielles 1998–1999, Centre de Mathématiques, École Polytechnique, Palaiseau, France, 1999, Exp. II. [Boutet de Monvel 3 (1999)] L. Boutet de Monvel, Complex star algebras, Math. Phys. Anal. Geom., 2-2 (1999), 113–139. [Boutet de Monvel 4 (1985)] L. Boutet de Monvel, Toeplitz operators: An asymptotic quantization of symplectic cones, in Stochastic Processes and Their Applications in Mathematics and Physics (Bielefeld, 1985), Mathematics and Its Applications, Vol. 61, Kluwer Academic Publishers, Dordrecht, the Netherlands, 1990, 95–106. [Boutet de Monvel 5 (2002)] L. Boutet de Monvel, Related semi-classical and Toeplitz algebras, in Deformation Quantization (Strasbourg, 2001), IRMA Lectures in Mathematics and Theoretical Physics, Vol. 1, de Gruyter, Berlin, 2002, 163–190. [Boutet de Monvel–Guillemin (1981)] L. Boutet de Monvel and V. Guillemin, The Spectral Theory of Toeplitz Operators, Annals of Mathematics Studies, Vol. 99, Princeton University Press, Princeton, NJ, 1981. [Boutet de Monvel–Sjöstrand (1976)] L. Boutet de Monvel and J. Sjöstrand, Sur la singularité des noyaux de Bergman et de Szegö, Astérisque, 34–35 (1976), 123–164. [Bouzouina–de Biévre (1996)] A. Bouzouina and S. De Biévre, Equipartition of the eigenfunctions of quantized ergodic maps on the torus, Comm. Math. Phys., 178-1 (1996), 83–105. [Cattaneo–Felder (2000)] A. Cattaneo and G. Felder, A path integral apporach to the Kontsevich quantization formula, Comm. Math. Phys., 212 (2000), 91–611. [Charles (2003)] L. Charles, Berezin-Toeplitz operators, a semi-classical approach, Comm. Math. Phys., 239-1–2 (2003), 1–28. [Connes (1974)] A. Connes, Non-Commutative Geometry, Academic Press, New York, 1994. [Delin (1998)] H. Delin, Pointwise estimates for the weighted Bergman projection kernel in Cn , using a weighted L2 estimate for the ∂¯ equation, Ann. Inst. Fourier (Grenoble), 48 (1998), 967–997. [de Biévre–degli Esposti (1998)] S. De Biévre and H. Degli Esposti, Egorov theorems and equidistribution of eigenfunctions for the quantized sawtooth and baker maps, Ann. Inst. H. Poincaré Phys. Th’eoret., 69-1 (1998), 1–30. [degli Esposti–Graffi–Isola (1995)] M. Degli Esposti, S. Graffi, and S. Isola, Classical limit of the quantized hyperbolic toral automorphisms, Comm. Math. Phys., 167-3 (1995), 471–507. [Dimassi–Sjöstrand (1999)] M. Dimassi and J. Sjöstrand, Spectral Asymptotics in the SemiClassical Limit, London Math Society Lecture Notes, Vol. 268, Cambridge University Press, Cambridge, UK, 1999. [Duistermaat–Singer (1976)] J. J. Duistermaat and I. M. Singer, Order preserving isomorphisms between algebras of pseudo-differential operators, Comm. Pure Appl. Math., XXVIV (1976), 39–47.


653

[Duistermaat–Singer (1975)] J. J. Duistermaat and I. M. Singer, Isomorphismes entres algebres d’operateurs pseudo-differentiels, in Seminaire Goulauoic-Lions-Schwartz Expose XXIV, Centre de Mathématiques, École Polytechnique, Palaiseau, France, 1975. [Etingof–Kazhdan (1996)] P. Etingof and D. Kazhdan, Quantization of Lie bi-algebras I, Selecta Math. (N.S.), 2 (1996), 1–41. [Gromov–Henkin–Shubin (1998)] M. Gromov, G. Henkin, and M. Shubin, Holomorphic L2 functions on coverings of pseudoconvex manifolds, Geom. Functional Anal., 8-3 (1998), 552–585 [Guillemin (1995)] V. Guillemin, Star products on compact pre-quantizable symplectic manifolds, Lett. Math. Phys., 35 (1995), 85–89. [Guillemin–Sternberg (1977)] V. Guillemin and S. Sternberg, Geometric Asymptotics, Mathematical Surveys, Vol. 14, American Mathematical Society, Providence, RI, 1977. [Hannay–Berry (1980)] J. H. Hannay and M. V. Berry, Quantization of linear maps on a torusFresnel diffraction by a periodic grating, Phys. D, 1-3 (1980), 267–290. [Helton (1977)] J. W. Helton, An operator algebra approach to partial differential equations: Propagation of singularities and spectral theory, Indiana Univ. Math. J., 26-6 (1977), 997–1018. [Howe (1980)] R. Howe, Quantum mechanics and partial differential equations, J. Functional Anal., 38-2 (1980), 188–254. [Karabegov–Schlichenmaier (2001)] A. V. Karabegov and M. Schlichenmaier, Identification of Berezin-Toeplitz deformation quantization, J. Reine Angew. Math., 540 (2001), 49–76. [Keating (1991)] J. P. Keating, The cat maps: Quantum mechanics and classical motion, Nonlinearity, 4-2 (1991), 309–341. [Kontsevich (1997)] M. Kontsevich, Deformation quantization of Poisson manifolds, Lett. Math. Phys., 66 (2003), 157–216. [Kontsevich (2001)] M. Kontsevich, Deformation quantization of algebraic varieties, Lett. Math. Phys., 56-3 (2001) (EuroConference Moshé Flato 2000 (Dijon), Part III), 271– 294. [Marklof–Rudnick (2000)] J. Marklof and Z. Rudnick, Quantum unique ergodicity for parabolic maps, Geom. Functional Anal., 10-6 (2000), 1554–1578. [Narnhofer (1997)] H. Narnhofer, Ergodic properties of automorphisms on the rotation algebra, Rep. Math. Phys., 39-3 (1997), 387–406. [Nonnenmacher (2003)] S. Nonnenmacher, unpublished note, 2003. [Reshetikhin–Takhtajan (1999)] N. Reshetikhin and L. Takhtajan, Deformation quantization of Kähler manifolds, in L. D. Faddeev’s Seminar on Mathematical Physics, American Mathematical Society Translation Series 2, Vol. 201, American Mathematical Soceity, Providence, RI, 2000, 257–276; math.QA/9907171, 1999. [Schlichenmaier (1998)] M. Schlichenmaier, Berezin-Toeplitz quantization of compact Kähler manifolds, in Quantization, Coherent States, and Poisson Structures (Białowiez˙ a, 1995), Polish Scientific Publishers PWN, Warsaw, 1998, 101–115. [Schlichenmaier (1999)] M. Schlichenmaier, Deformation quantization of compact Kähler manifolds by Berezin-Toeplitz quantization, in G. Dito and D. Sternheimer, eds., Conférence Moshé Flato 1999: Quantization, Deformations, and Symmetries, Vol. II, 1999, Mathematical Physics Studies, Vol. 22, Kluwer Academic Publishers, Dordrecht, The Netherlands, 2000, 289–306. [Schlichenmaier (1999b)] M. Schlichenmaier, Berezin-Toeplitz quantization and Berezin transform, in S. Graffi and A. Martinez, eds,m Long Time Behaviour of Classical and Quantum Systems: Proceedings of the Bologna Aptex International Conference, Bologna, Italy 13–17 September 1999, Series on Concrete and Applicable Mathematics, Vol. 1, World Scientific, River Edge, NJ, 2001.

654

S. Zelditch

[Shiffman–Zelditch] B. Shiffman and S. Zelditch, work in progress. [Shiffman–Tate–Zelditch (2003)] B. Shiffman, T. Tate, and S. Zelditch, Harmonic analysis on toric varieties, in J. Bland, K.-T. Kim, and S. G. Krantz, eds., Explorations in Complex and Riemannian Geometry: A Volume Dedicated to Robert E. Greene, Contemporary Mathematics, Vol. 332, American Mathematical Society, Providence, RI, 2003, 267–286. [Tamarkin (1998)] D. Tamarkin, Another proof of the M. Kontsevich formality thoerem, 1998, math/9803025. [Weinstein–Xu (1998)] A. Weinstein and P. Xu, Hochschild cohomology and characteristic classes for star-products, in Geometry of Differential Equations, American Mathematical Society Translation Series 2, Vol. 186, American Mathematical Society, Providence, RI, 1998, 177–194. [Zelditch (1997)] S. Zelditch, Index and dynamics of quantized contact transformations, Ann. Inst. Fourier (Grenoble), 47 (1997), 305–363. [Zelditch (1998)] S. Zelditch, Szegö kernels and a theorem of Tian, Internat. Math. Res. Notices, 6 (1998), 317–331.

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