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SU(2) WZW D-branes and their non-commutative geometry from DBI action


Preprint typeset in JHEP style. - HYPER VERSION

SU(2) WZW D-branes and their noncommutative geometry
arXiv:hep-th/0003057v3 21 May 2000

from DBI action
Jacek Pawelczyk

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Sektion Physik, Universit¨t M¨nchen a u Theresienstrasse 37 80333 M¨nchen, Germany u and Institute of Theoretical Physics Warsaw University, Ho˙ a 69, PL-00-681 Warsaw, Poland z Jacek.Pawelczyk@fuw.edu.pl

Abstract: Using properties of the DBI action we ?nd D-branes on S 3 of the radius Q5 corresponding to the conjugacy classes of SU(2). The branes are stable due to nonzero 2-form NSNS background. In the limit of large Q5 the dynamics of branes is governed by the non-commutative Yang-Mills theory. The results partially overlap with those obtained in the recent paper hep-th/0003037.

Work supported in part by Polish State Committee for Scienti?c Research (KBN) under contract 2P 03 B03 715 (1998-2000) and the Alexander-von-Humboldt Foundation.
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Recently it has been discovered that in a special limit the dynamics of the matrix model is described by the non-commutative Yang-Mills theory [1]. This has sparked new interest in NCG for strings propagating in NSNS antisymmetric tensor ?eld background [2]. Introduction of D-branes has provided deeper understanding of the role of non-commutativity [3] and it has allowed to derive conditions under which NCG starts to play dominant role in the dynamics of strings. It has also led to new understanding of the connection between quantum groups and WZW models [6, 8]. These two papers have used the standard CFT language what is a drastic bound on possible applications. In particular it does not allow to analyze RR backgrounds so much studied in the context of Maldacena’s conjecture [4]. The purpose of this paper is to provide understanding of the results of [6, 8] in the more universal language then that of WZW models. The hope is that after taking this lesson one would be able to derive interesting results for more general string/Mtheory backgrounds. Thus we shall describe various branes on the background of SU(2) WZW model using the D-brane e?ective action (DBI action) only. We shall also show how the non-commutativity appears in this approach. Methods applied here are limited to the case of large level of the SU(2) WZW model what in gravity language means large radius of the S 3 . Let us recall some of the results of [6] and [8]. D-branes in the level k SU(2) WZW model are in one-to-one correspondence with special integer conjugacy classes ghg ?1 for some ?xed h [6]. There are k + 1 of them: two D-particles (h = ±1) and k ? 1 D2-branes corresponding to two-spheres. The n-th sphere passes through the point exp(iπnσ 3 /k) ∈ SU(2), n = 1...k ? 1. We must also stress that D3-branes and D1-branes are excluded from this list. For large k the 2-spheres are in fact so-called fuzzy spheres [15]. The example of string theory background which involves the level k SU(2) WZW model is the near horizon limit of the F1, NS5 system (see e.q. [5]). Below we write only the relevant terms ds2 /α′ = Q5 d?2 3 H N SN S /α′ = 2Q5 ?3 e2φ = const. (1)

where Q5 denotes the number of NS5-branes and it is equal to the level k of the SU(2) WZW model, ?3 is the volume element of the unit 3-sphere. The e?ective action of the D-branes is given by DBI expression SDBI = ?Tp e?φ ?det[(X ? G + 2πα′F + X ? B)ab ] (2)

Vol

In the following we shall discuss classical con?gurations of branes embedded in S 3 of (1). Before we start to analyze equation of motion resulting from (2) we state

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several assumptions we make which seems to be natural here. We require the string coupling constant to be small and Q5 to be large in which case (1) is the part of an exact string background as at this limit supergravity is the perfect description of string theory. Moreover D-branes can be described completely classically by the DBI action. We also assume that the higher order correction to the DBI action are negligible. We shall be interested here only in the S 3 part of the con?guration thus it is even irrelevant if we consider IIB (as above) or IIA string. Thus some of the arguments given in our paper could be easily generalized to branes embedded in a 10d manifold of the form S 3 × M 7 under the condition that the embeddings are of the product structure i.e. the induced metric, pull-back of B and F ?elds are of block diagonal form. Recall that D-branes are de?ned to be the ends of the open strings. The string couple to the external sources (gauge A and B ?eld) as follows exp[ i ( 2πα′ 2πα′ X ? A + X ? B)] (3)



Σ

The example of the WZW model shows that the above formula can not be well de?ned globally for topologically non-trivial A and B ?elds. It is known that for closed strings i ?Σ = 0 the proper formula is exp[ 2πα′ Σ X ? H)] for H being locally dB and X is an extension of X to a 3-manifold Σ such that ? Σ = Σ. Now we consider con?guration of D-brane embedded into submanifold MD of the target space manifold M. One must repeat the above construction for the open string case [6, 7]. For the world sheet with one boundary the appropriate 3-manifold must respect ? Σ = Σ + D 2 . Rewriting the WZW model with boundary we get the proper global form of (3) 1 exp i ? 2πα′ X ? (2πα′ F + B) + X ?H (4)

D2

Σ

where X is an extension of X(?Σ) to a full 2-disc D 2 such that X(D 2 ) ? MD (F = 0 only on the D-brane manifold MD ). We stress that (4) has proper gauge invariance and for topologically trivial H it reduces to exp i ? 2πα′ X ? (2πα′ F ) + X ?B (5)

D2

Σ

i.e. to (3). Notice that one must be able to de?ne B on any X(D 2 ) thus we must have [H]MD = 0. The value of the integral (4) should not depend on the way one make the extension. This forces to put i 2πα′
1

C2

(2πα′ F + B) ?

i 2πα′

C3

H = 2iπm

(6)

? in front of the ?rst term is due to di?erent orientation of boundary ??Σ = ?D2 in D2 compare to Σ.

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where C 2 ∈ H2 (MD ) and C 3 ∈ H3 (M, MD ). Here a note is necessary concerning topology of the problem. For the argument we need an exact sequence of homologies . . . → H3 (MD ) → H3 (M) → H3 (M, MD ) → H2 (MD ) → H2 (M) → . . . (7)

If we assume that H3 (MD ) = H2 (M) = 0 then all cycles of H3 (M) are in H3 (M, MD ). i 3 Then one can write C 3 H = C 2 B mod 2π C 3 H = 2πQ5 m for CM ∈ H3 (M). Thus M the quantization condition reads
C2

F = 2πn,

n∈ Z

(8)

and n is de?ned modulo Q5 . This is the same as postulated in [12]. In the above we have disregarded the di?erence between the cycles in M and MD and their image given by X. D3 brane. Here we discuss the Dp-branes wrapped on the entire S 3 . According to the condition [H]MD = 0 we see that such a wrapping is impossible. We would like to provider here a di?erent argument based on DBI action. First one must notice that due to [H]MD = 0 the DBI action (2) is not well de?ned as B is not well de?ned on S 3 . In order to be more speci?c we concentrate on D3 brane in the background (1) and change the brane description to the dual form of the DBI action discussed e.g. in [10]. It has the same classical solutions as (2) what is the property we are interested in. ? ? (9) eφ ?det[(X ? G + 2πα′ F )ab ] ? πα′ F ∧ B SDBI ∝
Vol

The last term come form CS part of the DBI action. Integrating it by parts we get ? πα′ A ∧ H N SN S (10)

thus the action contains only the well de?ned B ?eld strength. With the H N SN S background given by (1) we see that there is a U(1) charge generated on the D3 world-volume. The charge can not stay on S 3 as it is a compact space, thus it forces the brane to partially unwrap the sphere. In the case of AdS3 ×S 3 the brane runs into the boundary of the AdS space. The above argument follows the baryon construction of [9]. D2 brane. Here we concentrate upon D2-brane case totally wrapped on S 3 . It can be also a e.g. partially wrapped D3 brane. We analyze its equation of motion and ?nd that contrary to the naive expectation the static brane it stable. As the indication of stability we invoke the lack of the tachyonic mode for the ?uctuation of the brane. In order to analyze the classical equations of motion we must ?nd out the pull back of B ?eld to the brane world-volume. On any 2-d submanifold of S 3 the B ?led is well (but not uniquely) de?ned. We have the freedom of changing B by an

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exact 2-form - in our case this will realized by choice of the solution for F12 . In the coordinates in which the metric on S 3 is ds2 = Q5 [dφ2 + sin2 (φ)d?2 ] we have for the 2 chart covering φ = 0 (11) B = Q5 α′ (φ ? ν ? 1 sin(2φ)) ?2 2 where ?2 is the volume form of the unit S 2 . We shall ?nd extrema of the DBI action corresponding to branes wrapped on S 2 given by some constant angle φ. The Euler-Lagrange equations are respected by 2πα′ F = ?Q5 α′ (φ ? ν) ?2 , φ(x) = φ = const. (12)

with all the other components of F equals zero. We also set ν = 0 requiring that the charge and the tension of the φ = 0 brane be zero. It is worth to note that the classical solution exists for any angle φ. When we apply the quantization condition (8) we get Q5 φ = 2πn (13) We remind that n is de?ned only modulo Q5 . We can compare (13) with results one gets assuming that the brane couple to some RR ?elds i.e. carry RR charge +Tp e2πα F +X
′ ?B


q

Cq

(14)

where, TDp = 1/((2π)p α′(p+1)/2 gs ). The background 2πα′F + X ? B generates RR charge of the D(p-2)-brane equals to Tp
S2 1 (2πα′ F + X ? B) = ?Tp (4πα′Q5 ) 2 sin(2φ).

One expects that this charge is integer multiple of T(p?2) i.e. 1 (2πα′F + X ? B) = ?2π n (15) 2πα′ S 2 but this is in contradiction with (13) for ?nite Q5 . If one takes the Q5 → ∞ limit then both formulae agree. 2 The second derivative of the DBI action with respect to the gauge ?elds and φ(x) gives kinematics of ?uctuations. One easily ?nds that ?uctuations of φ(x) only are massive but φ(x) mixes with gauge ?eld F leading to some massless modes [12]. Thus there is no tachyon in the spectrum and the brane con?guration is stable. Non-commutative geometry. We can also claim that at the Q5 → ∞ limit some of the branes are described by the non-commutative geometry. Here we follow the route of [3]. First we notice that at the Q5 → ∞ limit we have (nπ)2 2 d?2 → 0 Q5 2πα′ F + X ? B = ?α′ (nπ) ?2 ds2 = α′
2

(16)

The gap between (13) and (15) has been ?lled recently in [13].

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Thus the closed string metric goes to zero while induced 2πα′ F + X ? B is constant on the D2-branes world-volume what is a good sign for the non-commutativity. Next we calculate the open string metric and the Poisson structure inverting 2πα′ F + X ? (B + g). The inverse matrix is 1 + B) + 2πα′F = 1 Q5 sin φα′ sin φ cos φ ? cos φ sin φ (17)

X ? (g

Inverse of its symmetric part is the open string metric. We have Gab = α′ Q5 δab . Hence from the open string point of view all spheres have the same area! This, of course, is directly related to the ?at direction φ = const in the solution (12). The Poisson structure on S 2 (also called deformation parameter) is Θ12 = 2π 2 cot φ → Q5 n (18)

The symplectic structure is the inverse of the Poisson structure and it is ω12 = (n/2). One can check that this parameter precisely corresponds to the symplectic structure used by Berezin in order to quantize S 2 [14]. The non-commutative version on this S 2 is called the fuzzy spheres [15]. From [16] one may claim that the Y-M theory on this sphere is a theory of (n + 1) × (n + 1) hermitian matrices. Such a Y-M theory has (n + 1)2 degrees of freedom. Here we must stress that these results are in full agreement with [8]. It would be interesting to make explicit comparison of the brane dynamics and the above matrix model. We conclude that the branes dynamics is described by the non-commutative Y-M theory. The branes world-volume are 2-spheres which are non-commutative mani2 folds with the non-commutativity parameter Θ12 = n . A note added. Some of the results of this paper have been independently obtained in the recent paper [12].

Acknowledgments
I am grateful S.Theisen for illuminating discussions and reading the manuscript. I also thank K.Gaw?dzki, A.Alekseev, G. Arutyunov and A. Recknagel for comments e and interest in this work.

References
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[2] Y.-K.E. Cheung, M. Krogh, Nucl. Phys. B528 (1998) 185, hep-th/9803031 F. Ardalan, H. Arfaei, M.M. Sheikh-Jabbari, JHEP 9902 (1999) 016, hep-th/9810072 H. Garc? ?a-Compe?n, Nucl. Phys. B541 (1999) 651, hep-th/9804188; C. Chu and P. a Ho, Nucl. Phys. B 550 (1999) 151, hep-th/9812219 ; V. Schomerus, JHEP 9906 (1999) 030, hep-th/9903205 [3] N. Seiberg, E. Witten, hep-th/9908142. [4] J. M. Maldacena, Adv. Theor. Math. Phys. 2 (1998) 231, hep-th/9711200; S. S. Gubser, I. R. Klebanov and A. M. Polyakov, Phys. Lett. B 428 (1998) 105, hep-th/9802109; E. Witten, Adv. Theor. Math. Phys. 2 (1998) 253, hep-th/9802150 [5] J. Maldacena, A. Strominger, JHEP 9812 (1998) 005, hep-th/9804085 [6] A. Yu. Alekseev, V. Schomerus, Phys. Rev. D 60 (1999) 061901, hep-th/9812193. [7] K. Gawedzki, hep-th/9904145 ? [8] A. Yu. Alekseev, A. Recknagel, V. Schomerus, hep-th/9908040. [9] E. Witten, JHEP 9807 (1998) 006, hep-th/9805112. [10] C. Schmidhuber, Nucl. Phys. B 467 (1996) 146, hep-th/9601003; A.A. Tseytlin, Nucl. Phys. B 469 (1996) 51, hep-th/9602064. [11] D.S.Freed, E. Witten, hep-th/9907189. [12] C. Bachas, M. Douglas, C. Schweigert, Flux Stabilization of D-branes, hep-th/0003037. [13] W. Taylor, “D2-branes in B ?elds”, hep-th/0004141. [14] F.A.Berezin, Comm. Math. Phys. 40 (1975) 153. [15] J.Madore, Class.Quant.Grav.9 (1992) 69 [16] H. Grosse, C. Klimcik, P. Presnajder, Int. J. Mod. Phys. A 35 (1996) 231, hepth/9505175.

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