Scholarly article on topic 'T-duality of α′-correction to DBI action at all orders of gauge field'

T-duality of α′-correction to DBI action at all orders of gauge field Academic research paper on "Physical sciences"

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Abstract of research paper on Physical sciences, author of scientific article — Mohammad R. Garousi

Abstract By explicit calculations of four-field couplings, we observe that the higher derivative corrections to the DBI action in flat space–time, can be either in a covariant form or in a T-duality invariant form. The two forms are related by a non-covariant field redefinition. Using this observation, we then propose a non-covariant but T-duality invariant action which includes all orders of massless fields and has two extra derivatives with respect to the DBI action.

Academic research paper on topic "T-duality of α′-correction to DBI action at all orders of gauge field"

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Nuclear Physics B 909 (2016) 1-13

www.elsevier.com/locate/nuclphysb

T-duality of a '-correction to DBI action at all orders

of gauge field

Mohammad R. Garousi

Department of Physics, Ferdowsi University of Mashhad, P.O. Box 1436, Mashhad, Iran Received 15 March 2016; received in revised form 22 April 2016; accepted 24 April 2016 Available online 27 April 2016 Editor: Stephan Stieberger

Abstract

By explicit calculations of four-field couplings, we observe that the higher derivative corrections to the DBI action in flat space-time, can be either in a covariant form or in a T-duality invariant form. The two forms are related by a non-covariant field redefinition. Using this observation, we then propose a non-covariant but T-duality invariant action which includes all orders of massless fields and has two extra derivatives with respect to the DBI action.

© 2016 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license (http://creativecommons.org/licenses/by/4.0/). Funded by SCOAP3.

1. Introduction

The effective action of a Dp -brane in bosonic string theory includes various world-volume couplings of open string tachyon, transverse scalar fields, gauge field, closed string tachyon, graviton, dilaton and B-field. Because of the tachyons, the bosonic string theory and its Dp -branes are all unstable. Assuming the tachyons are frozen at the top of their corresponding tachyon potentials, the effective action at the leading order of a' in flat spacetime is then given by Dirac-Born-Infeld (DBI) action [1,2]

Sp d-Tpj dp+1aj- det(Gab + Fab) (1)

E-mail address: garousi@um.ac.ir. http://dx.doi.Org/10.1016/j.nuclphysb.2016.04.039

0550-3213/© 2016 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license (http://creativecommons.Org/licenses/by/4.0/). Funded by SCOAP3.

where Gab is pull-back of the bulk flat metric onto the world-volume,1 i.e.,

~ dxvdxv

Gab = P [T]\ab = daa dobnW

= nab + daX'dbXjntj (2)

where in the second line the pull-back is in static gauge,2 i.e., X1 = x' and Xa = oa. The DBI action (1) is covariant under the general coordinate transformations and is invariant under T-duality.3 With our normalization for the gauge field, the DBI action is at the leading order of a'. The first correction to this action is at order a' in which we are interested in this paper. The a' corrections to Born-Infeld action which includes only gauge field, have been studied in [3-8]. Using the proposed connection between relativistic hydrodynamics and open string effective action [9,10], the a' corrections to the DBI action may be used for studying higher-derivative corrections in relativistic hydrodynamics.

At zero gauge field level, the general covariance requires the world-volume couplings at any order of a' consist of various contractions of the second fundamental form £2abv = Da dX and its covariant derivatives. By studying the disk-level S-matrix element of two graviton vertex operators at low energy, such couplings at order a' have been found in [11] to be

Sp D -Tp

f dp+1oj- det(Gab)

1 + 2 *

+ a'l„vGabGcd{Qab^cdV - QaSttbd^ (3)

where R = Gvv GaPRvavp and Gvv is the first fundamental form, i.e.,

~liv dxv dxv ~ah

Gvv =--Gab (4)

doa do

which is a projection operator, i.e., nvaG^vGa^ = . It projects space-time tensors to the world-volume space. The tensor G^v in (3) is a projection operator, i.e., nvaGvvGap = , which projects space-time tensors to the transverse space. This projection operator can be written in terms of the first fundamental form as

v = n^v G^v (5)

In flat spacetime and in the static gauge, the transverse component of the second fundamental form in (3) is

1 Our index convention is that the Greek letters (v, v, • • • ) are the indices of the space-time coordinates, the Latin letters (a, d, c, • • •) are the world-volume indices and the letters (i, j, k, • • •) are the normal bundle indices. The killing index in the reduction of 10-dimensional space-time to 9-dimensional space-time is y.

2 In the literature, there is a factor of 2na' in front of gauge field strength Fab in the DBI action. We normalize the gauge field to absorb this factor. With this normalization, the gauge field along the killing direction, Ay, transforms to the transverse scalar field xy under T-duality.

3 By invariance under T-duality, we mean after expanding the action to a specific order of field, the couplings at each order satisfy the T-duality constraint (26).

&ab = dadbX' - GabCdcX'

= dadbX1 -GijdadbXknjk

= GijdadbXj (6)

and its world-volume component Uabc is zero.

The covariant action (3) includes all orders of the transverse scalar fields. Its two-scalar couplings do not change the scalar propagator as expected from S-matrix elements. We have also checked that its four-scalar couplings are consistent with the disk-level S-matrix element of four gauge bosons in the bosonic string theory which was calculated several years ago [16] (see Appendix).

In this paper, we are interested in including the gauge field Aa into the action (3). To this end, one may consider all gauge invariant couplings with unknown coefficients and impose the consistency of the couplings with the corresponding S-matrix elements to constrain the coefficients. There are further constraints if one requires the couplings to be covariant under the general coordinate transformations and/or to be invariant under T-duality transformations. We shall show that unlike the DBI action (1), the higher covariant derivative corrections to this action is not invariant under T-duality. As a result, we have to constraint the higher derivative couplings to be consistent with the S-matrix elements and to be either covariant under the general coordinate transformations or to be invariant under the T-duality transformations. In the latter case, we propose a T-duality invariant action which includes all orders of the gauge field.

An outline of the paper is as follows: In the next section, using the consistency of the couplings in flat spacetime with the general coordinate transformations and with the S-matrix element of four gauge bosons, we construct a particular four-field couplings at order a'. We then show that the couplings are not consistent with the T-duality transformations. To construct a T-duality invariant action, in section 3, we propose a non-covariant extension for the pull-back metric which is invariant under T-duality when the metric is not along the killing direction. Moreover, we introduce new tensors which are the transformations of the above object under the T-duality when it is along the killing direction. Using these non-covariant objects, we then construct a T-duality invariant action at order a' which includes all orders of the gauge field and is consistent with the S-matrix element of four gauge bosons. In section 4, we discuss our results.

2. Covariant action

In this section we are going to find four-field couplings at order a' which are consistent with the S-matrix elements and are covariant under the general coordinate transformation. The latter condition requires the couplings to be constructed from the gauge field strength Fab, its covariant derivative, i.e.,

Da Fbc = da Fbc Gab Fdc Gac Fbd

= da Fbc - GdidadbXiFdc + Gd idadcX Fdb (7)

and the second fundamental form Uabl.

The couplings of two transverse scalars and two gauge fields may have structure FFQQ or DFDF. We extend the square root in (3) to the DBI action, i.e.,

yj-det(Gab) ^yj- det(Gab + Fab)

Upon expand the square root, one finds a particular set of couplings with structure FFQQ. However, we have checked that they are not consistent with corresponding S-matrix element, i.e., they are not consistent with (38). As a result, the couplings may have other terms with structure FFQQ and/or couplings with structure DFDF. The latter couplings, however, should not change the propagator of gauge fields. So they must be total derivative at two-field level, i.e.,

Sp d -Tpj dp+1o^- det(Gab + Fab)

1 + a'I -DaFbcDaFbc + aDaFabDcFbcc

where the world-volume indices are raised by G"b and a is a constant. There are also 6 new couplings with structure FFQQ. The consistency with the S-matrix element, i.e., (38), can not uniquely fix the coefficients of these couplings. For example, if we do not consider the new couplings with structures FFŒŒ, then the S-matrix fixes a = 1.

To study four gauge field couplings at order a', one may consider all couplings with structure FFDFDF with unknown coefficients and constrains the coefficients by comparing them with the corresponding S-matrix element, i.e., comparing with (36). There are 18 such couplings and the comparison with (36) produces only three constraints. So three couplings are fixed and all others have unconstrained coefficients. One particular choice for the coefficients is

Sp d -Tpj dp+1aj - det( Gab + Fab) 1 + Q FaeFdeDaFbcDdFbc (10)

- 1 FceFdeDaFbcDaFbd - 1 FdeFdeDaFbcDaFb 3 6

The above couplings have been found in [5] by other means.

We have seen that there are many covariant couplings in (9) and (10) which are not fixed by the S-matrix element of four gauge bosons at order a'. Moreover, it is difficult to continue the above construction to find six-field couplings and higher orders. So one may use other consistency condition to fix the unknown coefficients at four-field level and possibly for higher orders. We are going to impose the constraint that like the DBI action (1), all higher derivative couplings to be invariant under the T-duality. However, the T-duality constraint is not consistent with the general covariance constraint when the higher derivative terms are included into the D-brane action. To see this point, we note that under T-duality Fab transforms to daxl when the gauge field is along the killing direction. On the other hand, while Fab appears at various places in (10), the velocity daxl appears only in the definition of the covariant derivative (7) and in the pull-back metric (2). In fact, we have considered all possible covariant couplings with unknown coefficients and constrained them to satisfy the T-duality invariance of the corresponding action. This produces a set of constraints which are not consistent with the constraints from the S-matrix elements. Therefore, the D-brane effective action at order O(a') which is consistent with the S-matrix elements and is invariant under T-duality may not be covariant under general coordinate transformations. In the next section we study the effective action which is invariant under T-duality transformation.

3. T-duality invariant action

The low energy expansion of an arbitrary S-matrix element can be separated into two parts. One part includes massless poles and the other part includes contact terms, i.e.,

A — Apole + ^contact (11)

The D-brane effective action must reproduce the contract terms in Acontact in the momentum space. On the other hand, it is known that the S-matrix element of an arbitrary number of gauge or transverse scalar vertex operators must satisfy the Ward identity corresponding to the T-duality [12,13]. Since the T-duality is a global duality, Apole and Acontact each must satisfy the Ward identity. In other words, the effective action must satisfy the linear T-duality after imposing the on-shell relations. Since the T-duality transformations on gauge and the scalar fields are linear, i.e., Ay ^ xy, the effective action must be consistent with an action which is invariant under the T-duality transformations. As we have observed in the previous section, the effective action, however, may not be in a covariant form under the general coordinate transformations.

Therefore, one should consider the non-covariant form for the couplings, i.e.,

dFdF + FFdFdF + FFFFdFdF + FFFFFFdFdF + ■■■ (12)

where dots represent higher order terms and the terms containing dx, ddx. The indices are contracted with flat metric.4 Each term has many different contractions. One should contribute an unknown constant for the coefficient of each contraction. One should then impose the condition that the action must be invariant under the T-duality. This constrains the coefficients. The resulting T-dual action must be also consistent with the S-matrix elements. This produces some further constraints on the coefficients.

Imposing the above two conditions, in principle, one can find four-field couplings, six-field couplings and so on. Since the T-duality is linear, there is no relation between these sets of T-dual couplings, e.g., the T-duality produces no relation between four-field couplings and six-field couplings. To find a relation between the above T-dual sets, we use an extra condition that the couplings should be consistent with all orders of scalar couplings in (3). To implement this latter condition, we propose to add appropriate gauge field into the pull-back metric and into the projection operator _LMV to make the couplings in (3) to be consistent with the T-duality. We begin by considering an extension for the pull-back metric to be consistent with T-duality.

When derivatives of the gauge field strength are zero, the T-duality may fix the presence of Fab in the inverse of the pull-back of the flat metric by extending it to the following expression:

/ 1 1 \ab

L_ab Gab — P[n] pr (14)

\P [n] + F P [n]-FJ

which is a symmetric matrix. To show that the above replacement is consistent with T-duality,

suppose the D-brane is along the circle on which the T-duality is imposed. When a, b are not the

killing index, i.e., a — a, b — b, using the prescription given in [15], one can verify that Gab is

invariant under T-duality. To the second order, it is

Gab — nab - daxldbxJmj + FacFdbncd

— nab - daxldbxinn + FacFdbncd - daAydbAynyy

4 One may also consider terms which contain the second derivative of gauge field strength and the third derivative of scalar fields, i.e.,

FFFddF + FFFFFddF + FFFFFFFddF + ■ ■ ■ (13)

However, such terms convert to the couplings in (12) by integration by part. So in the action we do not consider such couplings.

-U nab - daxdbx]m] + FacFdbncd - daxydbxynyy

= nab - daxldbxJmj + FacFdbncd = Gab (15)

We have checked it with the Mathematica to the tenth order and found that Gab is invariant. Inverse of the new metric (14) is

Gab = P Wab - FacFdbGcd (16)

which is not the pull-back of the flat metric in the static gauge, so the extension (14) does not have geometrical interpretation. As a result, an action which uses this matrix is not in a covariant form anymore. The matrix (14) defines a new form with space-time indices, i.e.,

„„ dxv dxv ab

G,x =---Gab (17)

3aa dab

We will find that all components of this form, i.e., Gab, Gai and Glj appear in the T-duality invariant action at order a'. Note that Gvv is not projection operator, so it is not a first fundamental form. This matrix has even number of gauge field strength.

When one or both indices of Gab are the killing index, it turns out that it transforms to the following expressions under T-duality:

Gya T > ®a y

Gyy -U ±yy (18)

Note that the y index on the left hand side is a world-volume index whereas on the right hand side it is a transverse index. The new matrix ±lj = nlj - Glj and matrix &ai is the following:

al ( 1 1 Yb i

&al = -F- dbxl (19)

\P [n] + F P M-FJ bx

We have checked the T-duality transformations (18) to the tenth order and found agreement. The presence of &al indicates that in a T-duality invariant theory there must be another tensor as

llv dXv dXv ab

=--j-&ab (20)

daa dab

where the new antisymmetric matrix &ab is

&ab i-1-F-1-^ (21)

Note that Gab - &ab is the inverse of the operator inside the square root in the DBI action (1),

ab ab ab

P [n] + F P [n]-F

jab _ Qab

i.e., (P~++Fyb = Gab - &ab. We will find that all components of (20), i.e., &ab, &al and &lj

appear in the effective action at order a'. Note that is not a projection operator. It has odd number of gauge field strength.

We have also found that &ab when a, b are not the killing index, is invariant under T-duality and found the following T-duality transformations:

®yi - Giy (22)

®ay T > Qa y

Gyi -U ®iy

which can be verified by expanding the matrices in both sides in terms of F and dx and using

the T-duality transformation Ay —> xy .

Therefore, in a manifestly T-duality invariant action there may be the matrices G^v, ®^v and 1ij which form a T-dual multiplet. Moreover, the action at order a' must include ddx and dF which form another multiplet. We are going to extend the scalar couplings in (3) to include the gauge field. This condition constrains the six indices of (ddx)2, ddxdF and (dF)2 to be contracted with six indices of GGG, GG1, GG® and so on. Taking the symmetries of these tensors, there are 41 different contractions.

Using the Mathematica package "xAct" [19], one can write all above contractions as

ClGad®be®cffabcfdef + C2Gad®bC®effabcfdef + C3GCd ®ae ®bf fabcfdef

+ C4GCd®ab®effabCfdef + cG ®ae ®bd fabcfdef + C6Gcf ®ad ®be fabcfdef + C7GCf®ab®defabcfdef + C&GaeGbd Gcf fabcfdef + C9Gad GbeGcf fabcfdef + CioGdf®ae®bCfabctdef + CllGdf®ab®Cefabcfdef + CUGabGCe Gdf fabcfdef

+ Ci3Gbd®aC®ijO,abiOJcdj + Ci4Gij®aC®bd^abi^cdj + Ci5GaCGbd Gij OlabiOJcdj + ci6GabGcdGijMabi^cdj + ci7lij®ac®bdo,abiOJcdj + c1&GacGbd 1ijO,abiOJcdj + Ci9GabGcd rivabiVcdj + C20®ai®be®CdUaeitbcd + C2® ®bd ®Ce Vdeifbac + C22®'"®bC®deVae1fbcd + C23GM GCe ®ai ^deifbac + C24GbC Gde ®ai ^aeifbcd

+ C25GbCGde®aiUdeifbac + C26GCd®ai ®bj^acj^bdi + C27GCd®ai ®bj^aci^bdj

+ C2&GCd®ai®bjUabiUcdj + C29GaiGM®CeO>aeifbcd + C3oGai Gbe®Cd^aeifbcd + C3lGalGbe®CdVdeifbac + C32Ga'GCe®bdVde,fabc + C33Gai GCe ®bd ^deifbac + C34GaiGde®bC0>aeifbcd + C3SGai Gde®bCOldeifabc + C36GaiGde®'CVdeifbac + C37Gbj®ai®CdUacjUbdi + C3&Gbj®ai®CdUaciUbdj + C39Gai Gbj GCd^acj^bdi + C4oGalGbjGcdVacl O^bdj + C41Gai Gbj GCdMabiMcdj — Lp (23)

where ci, ■ ••, c41 are unknown coefficients,

fabc = da Fbc, G>abi = da dbXi, (24)

and the contraction of indices in (23) are with the flat metric. Each term has even number of gauge field which is required by the invariance of the couplings under the parity. When expanding the matrices G^v, ®^v and 1ij around the flat metric, one finds a particular form for the series (12) which has only 41 unknown coefficients. The action which must be invariant under T-duality is

Sp — Tp

I dp+1aj- det(Gab + Fab)

1 + Lp + O(a')

where Lp is given in (23). Some of the couplings in (25) are total derivative terms that must be ignored and some other couplings are related to each other by the Bianchi identity. After

constraining (25) to satisfy the T-duality condition, we will remove the total derivative terms and impose the Bianchi identity to remove the couplings which are related by the Bianchi identity.

To constrain the couplings (25) to be consistent with the T-duality, following [15], we reduce the 10-dimensional space-time to the 9-dimensional space-time. It reduces (25) to two different actions Spw and S'p. In Spw, the killing direction y is a world-volume direction, i.e., a = (a, y) and in S'p the killing direction is a transverse direction, i = (i, y). The transformation of Spw under the T-duality which is called Sp^, may be equal to S'p_1 up to some total derivative terms which must be ignored in the action, i.e.,

SW_1 _ S'p _1 = 0 (26)

This constrains the unknown coefficients in the Lagrangian (23). Note that if one does not ignore the total derivative terms, then one would find some constraints which make the total derivative terms in the D-brane action to be T-duality invariant.

To impose the above constraint, one may expand the Lagrangian (23) around the flat metric. It is easy to verify that each term in (23) has contribution at the sixth order. So the T-duality rule (26) at order six, constrains all 41 coefficients. We expect there would be no further constraint at the eighth order and higher, because the higher order terms are resulted from expanding the matrices G'xv, and ±lj which are already shown to be connected under T-duality transformation to all orders.

We have expanded the Lagrangian (23) to the sixth order and imposed the T-duality constraint (26). We have found the following 23 relations between the constants:

C14 ^ 0,C15 ^ 0,C16 ^ 0,C22 ^ _2cio + C11 + 2c20,C23 ^ _C12 _ 2ci8 _ C19, C24 ^ 2c12 _ 2c17 _ C21,C25 ^ C12 _ C19,C26 ^ _C18,C27 ^ _C12 + 2c17 + C21, C28 ^ C12 _ 2C17 _ C19 _ C21,C29 ^ _2c10 + C11 + C12 + C19,

C32 ^ _3c12 _ 2c13 + 6c 17 _ 3c19 + 4c21 + C31,

C33 ^ C12 + 2C13 _ 2c 17 + C19 _ C21 _ C31,C36 ^ _2C10 + cn _ 2C35,

C37 ^ 2c12 _ 2C17 + 2C19 _ 2C21,C38 ^ _2C10 + C11 + C12 + C19,

C39 ^ _2c12 _ C13 + 3c17 _ 2c19 + 2c21,c40 ^ C30--—,

C41 ^ _2c10 + C11 + C12 + C19,

C5 ^ 2c 1 + C12 + C13 _ 3c 17 + C19 _ 2c21 _ C3,

C6 ^ _2c1 _ C12 _ C13 + 2c17 _ C19 + C21 + C3,

A , C34 , o c12 , c18 , c19 c8

C7 ^ _4C2 + C30 _ — + 2C4,C9 ^ — + — + — _ — (27)

After inserting the above relations on the coefficients in (23), one finds 18 T-dual multiplets. However, not all the coefficients of these multiplets are independent.

We have to impose on these 18 multiplets the condition that the couplings must be consistent with the scalar couplings in (3). This gives the following 5 constraints:

C13 3C17

C12 ^ _1 + 2c10 _ C11 ,C18 ^_1,C19 ^ 1,C21 ^ 2c10 _ C11 + —---—,

C34 ^ 2c30- (28)

We have to also impose the condition that the couplings must be consistent with the S-matrix element of four gauge bosons at low energy. We have already shown that the four-scalar couplings

in (3) are consistent with the corresponding terms in the S-matrix element, i.e., (37). So the above constraints include the consistency of the couplings with the S-matrix element of four scalars. The consistency of the couplings of four gauge fields with the corresponding terms in the string theory S-matrix element, i.e., (36), produces the following constraint:

ci7 ^ 3 + ci3 (29)

To find the above relation, we simply transformed the couplings to the momentum space and impose the on-shell relations and then compare them with the on-shell couplings in (36). With the above constraint, the couplings are also consistent with the S-matrix element of two gauge fields and two scalars.

So there are i3 T-dual multiplets in the action which are consistent with (3) and with the S-matrix element of four gauge bosons. There are 12 unknown coefficients in these 13 multiplets. These i2 coefficients are not independent yet. We now remove the couplings which are total derivatives and impose the Bianchi identity in the action. Writing the gauge field strength in daFbc in terms of gauge field, i.e., dadbA c — dadcAb, one finds the constants ci, c2, C3, C4, cg, c1o, c2o, c3o, c31, c35 do not appear in the action. That means the T-dual multiplets with these coefficients are zero by using the Bianchi identity. So it is safe to set all these 10 coefficients to zero. There are only two unknown coefficients c11 and c13 which appear in the following terms:

Tpcnj dp+1o^ — det(Gab + Fab)

— 2 GadGbeGcffabcfdef

— GabGceGdffabcfdef + Gcf®ae®bdfabcfdef + Gdf ®ab ®cefabcfde f

— GbcGde®alfbcdVaei + ®ai®bc®de^bcdVaei — GalGce®bdfabc^dei

+ GbdGce®a'^bac^de, — GbcGde®a'^bac^de, + Ga'Gde ®bc^bac^de,

— ®a'®bd®ce^bacVde

Tpc13 j dp+1ay — det(Gab + Fab)

— GbcGde®aifbcdO>aei + Gcd®ai®bjœa

'aci&bdj

- Gcd®ai®bj^abi^cdj + ±ij®aC®bdVabiVcdj + Gbd ®ac ®ij ^abi^cdj

+ Ga'Gce®bd^bacVde, - ®a'®bd®ce^baM (30)

The cn-terms are zero when gauge field is zero, whereas, the ci3-terms are zero when the scalar field is zero. We have expanded them to the sixth order and found that they are total derivative terms. So c11 and c13 can also be set to zero.

The final result which is invariant under T-duality, is consistent with the S-matrix element of four gauge bosons and reduces to (3) when gauge field is zero, is the following action:

Sp D —Tp

j dp+1a7 — det(Gab + Fab) 1 + GabGcd±ij^abi^cdj

— GacGbd ±ija>abiVcdj — 2 GadGbeGcffabcfdef — GabGceGdffabcfdef

2 8 + 3 Gf®-debet,bctdef — - GbGd^d.aei+ G'd®ai®^bdi

+ 3 Gbj®ai®CdVacjVbdi + 5 GCd®ai®bjVaciVbdj - 3 GCd ®ai ®bj ^abi^cdj 4

+ 31iJ®aC®bda,abiOJcdj + 2GbdGCe®aifbacOJdei - 2GbcGde®ai fbacVdei - 3GaiGCe®bdfbacadei - 2®ai®bd®cefbacadei\ + O(a'2)

When the transverse scalar fields are zero, only the terms in the second line are survived. They are consistent with the couplings found in [7,8]. The last term is exactly the one in [8], the sign of the first term is different because the sign of in [8] is different from the one in (3). The second term which is zero upon using the first order equation of motion, has not been considered in [8].

4. Discussion

In this paper, we have proposed an action to all orders of gauge field and transverse scalars which is invariant under T-duality, is consistent with all orders of scalar couplings known in the literature and is consistent with the S-matrix element of four gauge bosons. The action, however, is not covariant under the general coordinate transformations. On the other hand, if one imposes the condition that the action should be invariant under the general coordinate transformations and is consistent with the S-matrix elements, there are many unknown coefficients in the action even at the four field level. The general covariance and the S-matrix element constraints can not fix the coefficients of the couplings.

Since the T-duality transformations on the gauge field and on the transverse scalars are linear, the T-dual Ward identity of S-matrix elements indicates that the contact terms of the S-matrix elements of an arbitrary number of gauge bosons must satisfy on-shell T-duality relations. That means the couplings must be consistent with an action which is invariant under the T-duality transformation. On the other hand, the contact terms of the S-matrix elements must reproduce all orders of the scalar couplings in (3). That means the consistency of the couplings with all S-matrix elements indicates that the effective action may be invariant under the T-duality and at the same time be consistent with all scalar couplings in (3). If this constraint could not fix the coefficients of all couplings then one must impose other constraint, i.e., the consistency with the S-matrix element of gauge fields. Since the action (31) is consistent with T-duality, is consistent with all scalar couplings in (3) and has no unknown coefficients, we expect this action to be the effective action at order a' which includes all orders of gauge field. In other words, we expect this action to produce contact terms of all S-matrix elements. However, the field redefinition can change the form of action to many other forms. For example, a non-covariant field redefinition may change the form of action to covariant form. So we expect the action (31) to be unique up to field redefinitions.

We have found the result (31) by imposing the T-duality constraint (26) on the action, i.e., ignoring the T-duality constraint on total derivative terms. One may impose the T-duality constraint on the Lagrangian, i.e., C-1 - Ltp-1 — 0. To this end, we have used the T-duality transformations on G and ® that we have found in section 3. We have found the couplings in (31) and (30) with ci3 — -2/3 and cn — 0. So the T-duality constraint on the Lagrangian again produces the couplings (31) up to a total derivative term. In other words, the couplings (31) are invariant under T-duality to all orders of massless open string fields.

The B-field appears in the brane action in two different ways. Either through the different projections of its field strength H into world-volume and transverse space, or through the pull-back

of B-field P[B]. The latter, however, breaks the B-field gauge transformation unless it appears as the gauge invariant combination F + P[B]. So the gauge field strength in the action (31) should be extended as F ^ F + P[B]. However, this action is not in covariant form, so its extension to arbitrary metric gab is not simply to replace n ^ g and to change ordinary derivatives to covariant derivatives.

To include the gravity into (31), one may first expand the action around flat metric and use appropriate field redefinitions to rewrite the couplings in a covariant form, e.g., the couplings in section 2 for two and four gauge fields. Then one may extend the flat space metric into arbitrary metric by extending P [n] —> P [g] and extending the covariant derivatives (6) and (7) to include the derivatives of the metric. It would be interesting to find such covariant form for the action and see if there is a compact expression for the couplings which includes all gauge and scalar fields. The replacement F ^ F + P[B] in such covariant expression, then would produce many couplings between gravity and B-field.

The couplings between gravity and B-field should also appear through the scalar curvature [16,14]. It has been observed in [14] that the contact terms of the S-matrix element of two gravi-ton vertex operators in the presence of constant background B-field can be reproduced by the Riemann curvature contracted with Gab and ®ab. However, the metric in one of these matrices is flat metric. So the proposed couplings in [14] include all B-field but are not covariant as in the couplings in (31). We expect, in order to find the couplings in covariant form, one should expand the non-covariant form of the couplings found in [14] in a series in terms of B-field, and then look for a covariant action which reproduces the series. The result should include the covariant form of the couplings (31) in which F ^ B, as well as a series involving the couplings between B-field and the Riemann curvature.

The couplings between gravity and the transverse scalar fields at order a' are given in (3). In this paper, we have extended the transverse scalar couplings to include the gauge field strength by making the couplings in flat space-time to be consistent with T-duality. The consistency of the gravity part, for the special case of xi — 0, under linear T-duality has been used in [17] to find the dilaton and the couplings involving H — dB. It would be interesting to study the consistency of the action (3) which includes all scalar and gravity couplings at order a' under full nonlinear T-duality. The T-dual theory should then include all couplings of massless open and closed string fields at order a'.

We have seen that the couplings in (31) are consistent with the S-matrix element of four gauge bosons in flat spacetime. To verify that this action is consistent with the higher order S-matrix elements, one may consider the S-matrix element of four gauge bosons in the presence of background constant B-field. The replacement F ^ F + P [B] can produce such couplings in field theory. The disk-level S-matrix elements of four gauge bosons with mixed boundary condition in string theory, however, produce the couplings of non-commutative gauge fields [20,21]. So to produce such couplings from field theory (31), one should also use SW map [20] to transform the ordinary gauge fields in (31) to the non-commutative variables, and then compare them with the corresponding S-matrix element in string theory. We leave the details of such calculation to the future works.

The leading higher derivative corrections to the DBI action in the superstring theory are at order a'2. All transverse scalars corrections at order a'2 have been found in [18]. It would be interesting to apply the T-duality method used in section 3 to find the corrections which include all transverse scalars and gauge fields at order a'2.

Acknowledgement

This work is supported by Ferdowsi University of Mashhad under grant 2/39605(1394/11/04). Appendix A

In this appendix we find the low energy expansion of the S-matrix element of four gauge bosons in the bosonic string theory. The S-matrix element has been calculated in [16],

A1234 ---———- K' (32)

1234 r(1 + u) y ;

where the Mandelstam variables are s = -k1 k2, t = -k1 -k4, u = -k\-k3 which satisfies s +1 + u = 0, and K' is the following kinematic factor:

K' = -K + №1 -k3^2 ■k3(Z3 ■ kxZ4 ■ kx + Z3 ^4 ^2) 1

+ 3 (Z1 ^2 k - ■ k3Z2 ■ k1Z3 ■ k2)(Z4 ■ k1 - Z4 ■k2)] tu

+ --Z <2 - ■ k2Z2 ■ k1)(Z3 ■Z4 - Z3 ■ k4Z4 ^3) - tu^ ■ Z2Z3 ■ Z4}

+ {1, 2, 3,4}^{1, 3, 2, 4} + {1, 3, 2,4}^{2, 3, 1,4} (33)

where K is the kinematic factor of the corresponding superstring amplitude. It has four momenta and plays no role in the couplings of four gauge fields at the order of six momenta as we will see shortly. In above amplitude a' = 1 /2. Both K and K' are stu symmetric. The a'-expansion of the Gamma functions is

r(-s)r(-t) 1 n2 n4 2 2

'V ) ) = - - -r - Z(3)(s + t) - — (4s2 + st + 4t2) + ■ ■ ■ 1(1 + u) st 6 360

The total amplitude includes all non-cyclic permutations of the external states, i.e.,

A = A1234 + A1243 + A1324 + A1342 + A1423 + A1432 (34)

Using the relation s +1 + u = 0, one finds that A has no massless pole. It becomes

n2 + ^ (t2 + s2 + u2) + ■ •

K' (35)

It is clear now that the superstring kinematic factor K in K' has no contribution at six momenta in the total amplitude. It has contribution at four, eight, and higher momenta. The four momenta terms are reproduced by the DBI action (1) which are proportional to n2, and its eight momenta terms are reproduced by terms [18] which are proportional to n4.

The a'-expansion of the tachyon pole in K', produces the following on-shell couplings at six momenta which are proportional to n2:

Ast(A4) - {s[Z1 ■ k3Z2■ k3(Z3■ k1Z4■ k1 + Z3■ k2Z4^k2) 1

+ 3(Z1 ■ k2Z2■ k3Z3 ■ k1 - Z1 ■ k3Z2■ k1Z3 ■ k2)(Z4■ k1 - Z4■ k2)]

- tu(Z1 ■ Z2Z3 ■ k4Z4■ k3 + Z1 ■ k2Z2■ k1Z3 ■ Z4) - stuZ1 ^2Z3 ■ Z4}

+ {1, 2, 3, 4}^{1, 3, 2,4} + {1, 3, 2, 4} ^ {2, 3, 1, 4} (36)

The couplings for the transverse scalars can be found from the above couplings by using the condition that the scalar polarization is in transverse space, i.e., Zi • kj — 0. So the couplings for four scalars are

A6k(x 4) --stu(Z1 • Z2Z3 • Z4 + Z1 • Z3 Z2 • Z4 + Z1 • Z4Z2 • Z3) (37)

The couplings for two gauge fields with polarizations Z1, Z2 and two scalars with polarizations Z3, Z4 are

A6k(A2x2) ~-tu(Z1 • k2Z2• hZ3 • Z4) - stuZ1 •Z2Z3 • Z4 (38)

We compared the couplings (37) with four scalar couplings in (3) and found exact agreement. This fixes the normalization of the scatting amplitude (32). We compared the couplings (38) with two scalar and two gauge fields in (3) and (9) and found the unknown coefficient in (9) to be a — 1. The a'-expansion of the tachyon pole in K', produces also terms with eight, ten and higher momenta. All are proportional to n2. The terms with eight momenta may be reproduced by DUDU and its T-dual completion. Such terms are absent in the superstring theory.

References

[1] R.G. Leigh, Mod. Phys. Lett. A 4 (1989) 2767.

[2] C. Bachas, Phys. Lett. B 374 (1996) 37, arXiv:hep-th/9511043.

[3] A. Abouelsaood, C.G. Callan Jr., C.R. Nappi, S.A. Yost, Nucl. Phys. B 280 (1987) 599, http://dx.doi.org/10.1016/ 0550-3213(87)90164-7.

[4] A.A. Tseytlin, Phys. Lett. B 202 (1988) 81, http://dx.doi.org/10.1016/0370-2693(88)90857-X.

[5] O.D. Andreev, A.A. Tseytlin, Nucl. Phys. B 311 (1988) 205, http://dx.doi.org/10.1016/0550-3213(88)90148-4.

[6] N. Wyllard, Nucl. Phys. B 598 (2001) 247, http://dx.doi.org/10.1016/S0550-3213(00)00780-X, arXiv:hep-th/ 0008125.

[7] O. Andreev, Phys. Lett. B 513 (2001) 207, http://dx.doi.org/10.1016/S0370-2693(01)00676-1, arXiv:hep-th/ 0104061.

[8] N. Wyllard, J. High Energy Phys. 0108 (2001) 027, http://dx.doi.org/10.1088/1126-6708/2001/08/027, arXiv: hep-th/0107185.

[9] V. Niarchos, arXiv:1510.03438 [hep-th].

[10] G. Grignani, T. Harmark, A. Marini, M. Orselli, arXiv:1602.01640 [hep-th].

[11] S. Corley, D.A. Lowe, S. Ramgoolam, J. High Energy Phys. 0107 (2001) 030, arXiv:hep-th/0106067.

[12] M.R. Garousi, J. High Energy Phys. 1111 (2011) 016, http://dx.doi.org/10.1007/JHEP11(2011)016, arXiv:1106. 1714 [hep-th].

[13] K.B. Velni, M.R. Garousi, Nucl. Phys. B 869 (2013) 216, http://dx.doi.org/10.1016/j.nuclphysb.2013.01.001, arXiv:1204.4978 [hep-th].

[14] F. Ardalan, H. Arfaei, M.R. Garousi, A. Ghodsi, Int. J. Mod. Phys. A 18 (2003) 1051, arXiv:hep-th/0204117.

[15] M.R. Garousi, J. High Energy Phys. 1002 (2010) 002, arXiv:0911.0255 [hep-th].

[16] H. Kawai, D.C. Lewellen, S.H.H. Tye, Nucl. Phys. B 269 (1986) 1, http://dx.doi.org/10.1016/0550-3213(86) 90362-7.

[17] M.R. Garousi, A. Ghodsi, T. Houri, G. Jafari, J. High Energy Phys. 1310 (2013) 103, http://dx.doi.org/10.1007/ JHEP10(2013)103, arXiv:1308.4609 [hep-th].

[18] C.P. Bachas, P. Bain, M.B. Green, J. High Energy Phys. 9905 (1999) 011, arXiv:hep-th/9903210.

[19] T. Nutma, xTras: a field-theory inspired xAct package for Mathematica, arXiv:1308.3493 [cs.SC].

[20] N. Seiberg, E. Witten, J. High Energy Phys. 9909 (1999) 032, http://dx.doi.org/10.1088/1126-6708/1999/09/032, arXiv:hep-th/9908142.

[21] M.R. Garousi, Nucl. Phys. B 579 (2000) 209, http://dx.doi.org/10.1016/S0550-3213(99)00826-3, arXiv:hep-th/ 9909214.