T-dualization in a curved background in absence of a global symmetry 1

: We investigate T-duality of a closed string moving in a weakly curved background of the second order. A previously discussed weakly curved background consisted of a (cid:13)at metric and a linearly coordinate dependent Kalb-Ramond (cid:12)eld with an in(cid:12)nitesimal strength. The background here considered di(cid:11)ers from the above in a coordinate dependent metric of the second order. Consequently, the corresponding Ricci tensor is nonzero. As this background does not posses the global shift symmetry the generalized Buscher T-dualization procedure is not applicable to it. We rede(cid:12)ne it and make it applicable to backgrounds without the global symmetry.


Introduction
T-duality [1][2][3][4][5] was first introduced to represent the fact that the toroidal compactifications [6][7][8][9] of a closed string to a radius R and a radius 1/R are equivalent. Although the compactified theories are defined for different target spaces, their spectrum is the same. The observed symmetry lead to investigation for discovering the connections between the theories having the same spectrum, what resulted in T-dualization procedures. These prescriptions consist of rules which transform the given theory to its T-dual theory. The T-dual theories describing strings moving in a geometrically different backgrounds, having the same predictions, were found for some particular backgrounds. The general procedure, applicable to an arbitrary background is still to be determined.
T-duality was found to be connected with the isometries of a sigma model. This discovery was included as an inevitable condition for T-dualization, as the isometry was JHEP11(2015)119 built in the T-dualization procedure. The first procedure determining the T-duals of the constant background fields was the Buscher procedure [10][11][12][13]. This procedure, called the standard T-dualization procedure, is founded in localizing the global isometry by introducing the gauge fields, whose field strength is set to zero by a Lagrange multiplier term. The gauged theory reduces to the initial theory for the equations of motion for the Lagrange multiplier and to the T-dual theory for the equations of motion for the gauge fields. This procedure enabled investigation of the coordinate dependent backgrounds as well, when the T-dualizations are performed along the directions which do not appear as the background fields arguments.
The generalized T-dualization proposed in paper [14], addressing the non-abelian isometries lead to observation that the application of T-dualization procedures can lead to theories without an isometry. These theories are obviously T-dual to the initial theories, but, the initial theories can not be obtained as a result of the same T-dualization procedure starting with the theory without isometry. This observation implied that T-duality in general must be understood from some other perspective.
The investigation of the relations between non geometric backgrounds lead to a new generalized T-dualization in string field theory [15]. It was proposed that particular non geometric backgrounds should be understood as string backgrounds which are the result of generalized T-dualization applied along nonisometry directions. In paper [16], the conditions for a background to have a geometric or non geometric T-dual were sought for. It was concluded that the large class of sigma models that cannot be gauged can be T-dualized.
In paper [17], one considers similarity transformations of the stress energy tensor of a conformal field theory which do not change the Virasoro alebra. There exists the transformations of the background fields which produce the same change of the stress tensor as the change generated by some similarity transformations. A particular generator of a similarity transformation produces symmetry transformation, such as general coordinate transformations and gauge transformations of a Kalb-Ramond field. However, some particular forms of these generators produce T-duality transformations at critical radius. Investigation leads to T-dualization techniques directly applicable to an arbitrary string backgrounds.
In paper [18], a generalization of a Buscher T-dualization procedure was given. The generalized procedure is applicable to backgrounds depending on all the space-time coordinates, along arbitrary background fields argument. The procedure was realized for a weakly curved background which consists of a constant metric and a coordinate dependent Kalb-Ramond field with an infinitesimal strength. The difference between the generalized and standard Buscher procedure is in an invariant coordinate. Standardly, one substitutes the derivatives with the covariant derivatives to obtain the gauge invariant action, but in the generalized procedure one additionally substitutes the argument of the background field with the invariant argument. It was confirmed in [18] that the generalized T-dualization procedure does not harm the interchange of equations of motion and Bianchi identities [19]. However, it strongly changes the geometry of a target space. The geometric space is transformed to a double non-geometric space. The commutative space is transformed to a non-commutative space, as shown in [20]. The closed string non-commutativity was previously investigated in [21][22][23][24][25]. The application of a procedure to an arbitrary set JHEP11(2015)119 of coordinates was considered in [26]. It was concluded that the geometric background again transforms to a double space, with double coordinates present for both T-dualized and undualized directions.
In the present paper, we consider the weakly curved background of the second order. We take a metric which consists of a constant and quadratic in coordinate term and linearly coordinate dependent Kalb-Ramond field. This background does not posses the global shift symmetry. In comparison to the previously considered backgrounds there is an additional difference. The Ricci tensor of the metric here considered is nonzero. The background has to be the solution of the space-time equations of motion, obtained from the demand of the conformal invariance of the quantum theory. To satisfy these equations one takes the coordinate dependent parts to be infinitesimal.
The original form of the generalized Buscher T-dualization procedure [18] is not applicable to a weakly curved background of the second order. Here, we search for the procedure which will be applicable and will preserve the general features of the previous procedure. We find the appropriate formulation and investigate the properties and the consequences of the new generalization. We apply the procedure along all space-time coordinates and obtain the T-dual theory. We obtain a geometrical structure that differs from the double non geometrical space. The dual background field arguments do not depend only on the dual coordinate and its double. However the application of the procedure to all dual coordinates leads again to the initial theory. We obtain T-dual coordinate transformation laws and confirm that T-duality interchanges equations of motion and Bianchi identities.

Bosonic string action and choice of background
Let us consider the closed bosonic string propagating in the background fields: a metric G µν and a Kalb-Ramond antisymmetric tensor field B µν , described by the action The integration goes over two-dimensional world-sheet Σ parametrized by ξ α , α = 0, 1 (ξ 0 = τ , ξ 1 = σ). The coordinates of the D-dimensional space-time are marked by x µ (ξ), µ = 0, 1, . . . , D − 1. From the action principle one obtains the equations of motion is a Christoffel symbol. Introducing the light-cone coordinates and their derivatives the action (2.1) can be rewritten as

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where Π ±µν is the combination of background fields, defined by The equation of motion (2.2) can be rewritten as In order to obtain a conformally invariant quantum theory, the background fields must obey the space-time equations of motion, which for the constant dilaton field have the following form where R µν is Ricci tensor defined by and D µ is a covariant derivative (2.10) We will consider the following solution of the space-time equations of motion (2.7), (2.8) where B µνρ is constant and infinitesimal. Throughout the paper the calculation will be done up to the second order in B µνρ . We will refer to this solution as the weakly curved background of the second order. More general discussion about the solutions of the space-time equations of motion, up to the second order terms, can be found in ref. [27].
Let us demonstrate that (2.11) satisfies (2.7) and (2.8). The inverse metric and the Cristoffel symbol are which is just the eq. (2.7). The equation (2.8) is satisfied, because the term corresponding to the first term in (2.10) is zero and the others can be neglected as the third order terms in B µνρ . Let us notice, using (2.9) and (2.13), that the coefficient in the second order term of the metric (2.11) is in fact the Riemann curvature tensor

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The solutions which where previously investigated in this context where the constant background and the weakly curved background of the first order. In both cases the Ricci tensor R µν is absent, in the first case because it equals zero and in the second because it is neglected as the second order term. Here, the Ricci tensor is of the second order and its contribution becomes nontrivial because we work up to the second order in B µνρ .

T-dualization procedure
In the majority of papers addressing T-dualization of a bosonic string theory, one performs T-dualizations along directions on which the background does not depend. The first procedure, applicable to coordinates on which the background fields depend, the generalization of the Buscher T-dualization procedure, was presented in [18]. It was applied to a bosonic string moving in the weakly curved background, composed of a constant metric and a linearly coordinate dependent Kalb-Ramond field with an infinitesimal strength. This theory has a global shift symmetry. This fact is used in the T-dualization prescription, which relies on gauging the global symmetry. The locally invariant action was built substituting the ordinary derivatives with the covariant ones and substituting the coordinate in the argument of the background fields with the invariant coordinate (a line integral of a covariant derivatives of the original coordinates). The physical equivalence was achieved by introduction of the Lagrange multiplier term, which makes the gauge fields nonphysical.

Auxiliary action
Here, we will consider the weakly curved background of the second order. As in the first order weakly curved background, the Kalb-Ramond field is linear in coordinate and has an infinitesimal field strength. The metric however, beside of a constant term has a quadratic in coordinate part which is an infinitesimal of the second order. Such a metric has an infinitesimal but nonzero Ricci tensor R µν = 0. The bosonic string theory in this background does not possess the shift symmetry. However, defining of the new Tdualization rules on the grounds of the existing procedure is still possible. The main object in the conventional procedure, is the gauge fixed action which reduces to the initial action for the equations of motion for the Lagrange multipliers and becomes T-dual action for the equations of motion for the gauge fields. Here we will define its substitution, which inherits these two features. We postulate the auxiliary action by It can be obtained from the initial action (2.4), by making the following substitutions and adding the Lagrange multiplier y µ term. This action is of the same form as the gauge fixed action, however, v µ ± are here some auxiliary fields, which take over the role of the

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gauge fields. Similarly as in [18], the argument of the background fields is the line integral of the auxiliary fields taken along a path P (from ξ 0 to ξ) Note that as well as in ref. [18], the equation of motion with respect to y µ forces the "field strength" to vanish ∂ + v µ − −∂ − v µ + = 0, which is just the condition for the path independence of ∆V µ . In the resulting theories, the argument reduces to ∆V µ = V µ (ξ) − V µ (ξ 0 ) and we will chose the value of V µ (ξ 0 ) to be zero.

From the auxiliary to the initial and T-dual theory
Let us confirm that the auxiliary action (3.1) becomes the initial action (2.4) for the equations of motion obtained varying over the Lagrange multiplier y µ , and therefore taking x µ (ξ 0 ) = 0 the auxiliary action reduces to the initial action (2.4). The equations of motion for the auxiliary fields v µ ± are Here the functions β ± µ are defined by where δ V S aux stands for the variation of the action (3.1) over the background field argument V µ . Let us introduce the following background fields: an effective metric and a non-commutativity parameter, defined by and their combinations which are the inverses of the background field compositions 2κΠ ∓µν . Now, one can rewrite the equations of motion (3.6) as

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The equation (3.10) is not the solution of (3.6), because v µ ± appears within the argument V µ of both Θ µν ± and β ∓ µ . We will solve this equation iteratively. The T-dual theory is obtained, by inserting the equation of motion (3.10) into the action (3.1) In order to obtain the explicit form of the T-dual action one has to calculate the beta functions β ± µ for a concrete background, solve (3.10) to find the explicit y-dependence of the auxiliary fields v µ ± = v µ ± (y), and therefrom determine the argument of the dual background fields V µ (y).

T-dual action in a weakly curved background
Let us find the explicit expression for the T-dual action (3.11), in the weakly curved background of the second order. The main task is to obtain the β ± µ functions (B.6), which are calculated in appendix B. Because they are infinitesimal, it is enough to consider their first order value and to determine the zeroth order value of V µ , in order to calculate the last term in the action Let us find the explicit form of the dual background fields argument. We will solve the equations (3.10) iteratively and find the zeroth and the first order in B µνρ values of the auxiliary fields v µ ± (y). In the zeroth order one has consequently the zeroth order value of V µ defined in (3.3) is whereỹ µ is a double coordinate defined bỹ Now, using (4.3) and (A.8), the last term (4.1) in the T-dual action (3.11), becomes with ∆ µν ± explicitly given by (A.9).

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The first order value of the auxiliary field v µ ± , defined by (3.10), is obtained using the first order value of β ± µ , (B.6), and the expressions for Θ µν 1± given by ( Let us note that, because of (4.2) and (4.6), the complete first order value of the auxiliary field can be written as v where Θ µν ± is defined in (A.14). Substituting (4.6) into (3.3), we obtain the first order value of V µ and (y +ε . Once the argument of the background fields is calculated, we can write the explicit form of the T-dual action given by (4.3) and (4.8). The second term in the dual background fields composition ∆ µν − is the contribution from the term quadratic in β, and has a form (A.9).
Comparing the initial action (2.4) with the T-dual action (4.10), one can conclude that they are equal under the following transformations The T-dual metric (the symmetric part of the T-dual background fields composition) and the T-dual Kalb-Ramond field (the antisymmetric part) are

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and The characteristics of the dual geometry, are considered in section 7.

T-dual of T-dual
Let us now follow the prescription of section 3, and show that the T-dual of a T-dual theory is the original theory. To obtain the auxiliary action of the T-dual action (4.10), let us substitute the dual coordinate derivatives ∂ ± y µ with some auxiliary fields u ±µ , substitute the coordinate in the argument of background fields with ∆U µ = (dξ + u +µ + dξ − u −µ ) and require the "flatness" of u ±µ by introducing the Lagrange multiplier terms For the solution u ±µ = ∂ ± y µ of the equations of motion ∂ − u +µ + ∂ + u −µ = 0, which are obtained varying the auxiliary action over the Lagrange multiplier z µ , the variable U µ reduces to y µ (y µ (ξ 0 ) = 0). So, the auxiliary action reduces to the original one.
The original theory should be obtained for the equations of motion for the auxiliary fields u ±µ with β ∓µ defined by (C.2), being the contribution from the variation over the background fields argument. Multiplying the equations by † Π ∓µν (the inverse of the background field composition † Θ µν ± , defined in (A.11)) one obtains Using the last equation and the first order value of the dual beta function β ∓ν given by (C.15), we can determine the value of the variable U µ , up to the first order with M µν ± (z) defined in (4.9). Substituting (5.4) to (4.3) and (4.8) we confirm that V µ (U ) = z µ . So, substituting (5.3) to the action (5.1), we obtain Using the first order value of β ±µ , given by (C.15), the second term of the action becomes −2κ∂ + z µ (Π 0+ ∆ − (z)Π 0+ ) µν ∂ − z ν and therefore the action (5.5) is just the initial action (2.4)

JHEP11(2015)119 6 Features of T-duality
In the previous sections, we showed how the original and its T-dual theory can be transformed one to the other. In both directions, both theories follow from the auxiliary action and are obtained for a concrete form of the auxiliary fields. Comparing these auxiliary fields one obtains the T-dual coordinate transformation laws.
In section 3, we showed how the original theory can be transformed into its T-dual theory. So, comparing the expressions for the auxiliary fields (3.5) and (3.10), one obtains the T-dual coordinate transformation law In the first order this law implies Substituting the beta functions (B.6) into the transformation law (6.1), we obtain with Θ µν ± are ∆ µν ± given by (A.14) and (A.9). Using these laws one can show that the equation of motion of the original theory transform to an identity (Bianchi identity) in the T-dual theory, and vice verse. From (6.1) and (6.3), using (6.2) one obtains In section 5, the T-dual theory was transformed to the original theory. Comparing the solutions for the auxiliary fields we obtain the following T-dual coordinate transformation law κ∂ ± y µ ∼ = −2κ † Π ∓µν (z) ∂ ± z ν ± κ β ∓ν (z) . (6.5) In the first order this law implies Substituting the explicit value of the dual beta function (C.15), we obtain with Π ∓µν defined in (A.15). Eliminating ∂ ± z µ from (6.5) and (6.7), using (6.2) one obtains Let us show that the T-dual coordinate transformation laws (6.1) and (6.5) are inverse to each other. Multiplying (6.5) by † Θ ± (V (y)) ∼ = † Θ ± (z) we obtain κ † Θ µν ± (V (y))∂ ± y ν ∼ = −∂ ± z µ ∓ κ β ∓µ (z). (6.9)

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Using (C.15), (A.10) and (A.14) it becomes Recalling the definitions (A.9), (A.8) and (B.6) the last two terms cancel out and one obtains which is just (6.1). The equivalent conclusion that (6.3) and (6.7) are inverse to each other, follows from (A. 16). Let us finally show, that using the T-dual coordinate transformation laws one can confirm that the equations of motion and the Bianchi identities of the original and T-dual theory interchange. Applying the transformation law (6.7) to the identity we obtain Using the explicit form of the composition Π ±µν , given by (A.15), expression (A. 19) and the value of the Christoffel symbol (2.13), we obtain (6.14) So, (6.13) is the initial equation of motion (2.6).
The equation of motion of the T-dual theory (4.10) is Using the T-dual coordinate transformation law (6.7) (with z µ = x µ ) and (6.2), we obtain which with a help of (A.16) is just the identity

Original and dual geometries
Let us discuss what the geometry of the T-dual theory looks like and compare it with the geometry of the original theory. To simplify discussion we will put the constant part of the original Kalb-Ramond field, b µν , to zero. In fact it appears in front of a topological term and can contribute only in the quantum theory.

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Let us first note the substantial difference between our T-dual theories and the standard σ-formulations of string theories. In our approach argument of the background fields is expression V µ , which is a line integral of the T-dual coordinate derivatives. For b µν = 0 it essentially depends on a double coordinateỹ µ ≡ P dξ α ε β α ∂ β y µ , eq. (4.4), which makes the T-dual theory non-geometric. In some particular examples such theories are known as the theories with R-flux. For these theories, the equations of motion are not necessarily equal to the standardly derived space-time equations of motion for the background fields depending just on the coordinate x µ or y µ . Although we do not expect that all relations between background fields of the original and T-dual theories in our approach will coincide with those in the literature, we are going to compare them.
Let us first make a simple qualitative analysis. In the approximation of the first order it is easy to see, without calculation, that the T-dual space-time equations of motion are satisfied. In fact both dual metric G µν and dual Kalb-Ramond field B µν are linear in coordinates with infinitesimal coefficients. Consequently, the dual Christoffel Γ νρ µ and the dual field strength B µνρ are constant and infinitesimal. So, both dual space-time equations, for the metric and for the Kalb-Ramond field, are equal to the second order infinitesimals which are neglected, meaning they are satisfied. In our case of the second order approximation, a similar analysis shows that both Riemann tensor and square of the Kalb-Ramond field are constant and the second order infinitesimals in both initial and T-dual theories.
In this section we are going to discuss the following issues: the geometries and the space-time equations of motion of the initial and T-dual theories as well as the integrability conditions of ref. [28].

Geometry of the original theory
For the original theory we take so that the corresponding Christoffel symbols are linear in coordinate and infinitesimals of the second order while the Kalb-Ramond field strength is a constant infinitesimal of the first order Therefore, the Riemann tensor is a constant infinitesimal of the second order which produces the constant second order infinitesimal Ricci tensor Note that the covariant derivative of the field strength is equal to the ordinary derivative D µ H µ ρσ = ∂ µ H µ ρσ . This is the consequence of the fact that the Christoffel symbols are

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infinitesimals of the second order and the terms ΓH are infinitesimals of the third order which should be neglect in our case. When H µ ρσ is constant one has D µ H µ ρσ = 0. Therefore, the space-time equations of motion can be written in the form where for future benefits, following ref. [28], we introduced the tensors and Note that the coefficients in front of the squares of field strength differ from that in ref. [28], because of a different notation. In both articles they are adjusted in such a way that S µν = 0 is the space-time equation of motion.

Geometry of the T-dual theory
The background fields of the T-dual theory are In comparison to the original theory, the term h 2 of the metric tensor is missing and the background fields depend on V µ instead of x µ . The dual metric is constant and therefore the dual Christoffel symbol, dual Riemann and Ricci tensors are zero. But, the dual Kalb-Ramond field strength is constant infinitesimal of the first order H µνρ = −B µνρ . As we explained in the beginning of this section the T-dual fields do not satisfy the standard space-time equations of motion because the space is nongeometric and the background fields depend on the dual coordinateỹ. The T-dual space-time equations of motion are where again dual covariant derivative is equal to the ordinary derivative. It is interesting to note that although the initial theory is curved, the corresponding T-dual is flat. It seems that at least in the second order the T-duality acts as a parallelizable transformation. This assumption should be checked in the higher orders of approximations.

Relation with ref. [28]
Although, as we explained, we should not expect for our background to satisfy the pseudoduality conditions of ref. [28], we are going to discuss the relation with this article. Let us

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first note that β ± µ functions, introduced in the generalized T-dualization procedure, originate from the fact that T-dual background fields do not depend on the coordinate y µ but on its dual V µ = (g −1 ) µνỹ ν . So, in order to compare our relations with the conditions derived in the literature we will omit the term β − µ Θ µν − β + ν . Then, the T-dual metric tensor acquires the quadratic term and the Kalb-Ramond field is unchanged Secondly, one can note that the pseudoduality relation in ref. [28], which is the starting point in that paper corresponds to the relation (6.7) in this paper. Taking b µν = 0 the relation (6.7) reduces to where T ± is the notation from the article [28] where only the case T + = T − was treated. Obviously, the T-dual coordinate transformation laws differ at least by the term 3h. The Christoffel symbol and the Kalb-Ramond field strength for the background fields (7.11) are The Riemann tensor is 14) and the Ricci tensor equals Note that the Christoffel symbols, Riemann and Ricci tensors are one third of the corresponding variables of the original theory. The same as in the original theory, the Christoffel symbols are infinitesimals of the second order and the covariant derivative of the field strength is equal to the ordinary derivative D µ H µρσ = ∂ µ H µρσ . Because the tensor H µρσ is constant the right hand side is zero.
The dual space-time equations of motion can be written as where we define dual tensors S ρ σµν with additional coefficient 1 3 in the last three terms in comparison to the tensor S ρ

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The pseudoduality conditions of the ref. [28], in our notation read as follows Note that because both equations are infinitesimal we can raise and lower indices with the constant part of the metric. Both pseudoduality conditions are fulfilled because all terms are separately equal to zero. The second relation is valid without derivatives as well H µ ρσ = −H µ ρσ .

Conclusion
In this paper, we presented the T-dualization procedure applicable to string backgrounds with nontrivial Ricci tensor and without isometries. The procedure is the generalization of the one given in paper [18], for a weakly curved background. It was applied to a string moving in the weakly curved background of the second order, composed of a linearly coordinate dependent Kalb-Ramond field with an infinitesimal strength and a metric with an infinitesimal of the second order quadratic in coordinate term. The generalized Buscher procedure was not applicable to the second order weakly curved background, because the action does not possess a global symmetry. If there is no global symmetry, there is no corresponding gauge symmetry, which is the crucial ingredient of the T-dualization procedure. However, it is possible to construct an auxiliary action, which plays the role of the gauge fixed action. The auxiliary action is constructed from the initial action, substituting the derivatives of the coordinates by some auxiliary fields, and the background fields argument by a line integral of these auxiliary fields. This action reduces to the initial action and to the T-daul action on its equations of motion. So, there is a full analogy between the T-dualization procedures for backgrounds with and without a global symmetry. The only difference is in fact the interpretation of the auxiliary fields which are understood as the gauge fields in the case of a background with symmetry.
The realization of the new generalized Buscher procedure is more complicated. The main problem is to solve the equations of motion, obtained varying the auxiliary action with respect to the auxiliary fields, in terms of the Lagrange multipliers. To solve them, one should iteratively calculate the argument of the background fields and the beta functions defined in appendices B and C. It turns out that the argument of the dual background fields has a more complicated form then in the weakly curved background of the first order. This argument represents the complicated structure of the dual geometry. In the first order the argument is given in terms of the dual coordinate y µ and its doubleỹ µ . In the second order the argument is given in terms of the dual coordinate, its double and an additional form ±µ , which can be interpreted as the left and the right "angular momentum".
Applying the T-dualization procedure to all the coordinates of the initial theory, the theory transforms to a T-dual theory. The initial background which is curved and geometric transforms to a non geometric curved background

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where Θ µν − is defined in (4.11). Consequently the T-dual theory can not be directly compared with the standard theories, where the background fields depend on the ordinary coordinates. The T-dual Riemann tensor is zero, which means that T-dual background is flat. It would be interesting to check whether T-duality in the higher orders can make the target space parallelizable. Although the T-dual background is flat, certain adjustments can be made in order for our approximation to satisfy the relations analogue to the general relations of ref. [28].
Applying the procedure to all the dual coordinates, T-dual theory transforms to the initial theory. Comparing the solutions for the auxiliary fields we obtain the T-dual coordinate transformation laws, connecting initial and dual coordinates, which are inverse to each other. Using these laws one confirms that the equations of motion and the Bianchi identity of one theory transform to the Bianchi identity and the equations of motion of the other theory. Because these laws have obtained the second order correction, they will enable further investigation of the non-commutativity properties of the spaces connected by T-duality. Furthermore, the laws are the basis for a double formulation [29][30][31][32] where T-duality is interpreted as an exchange of the initial and dual coordinates.
So, we showed that the T-dualization of the theory with a non-trivial Ricci tensor and without global symmetry is possible, and that it does not break the standard features of T-duality. The non geometric structure of T-dual theory is much richer than in the cases previously analyzed and may be a subject of further investigations.

A The expansion of the background fields
All the expressions will be divided into its zeroth, first and second order values, for example G µν = G 0µν + G 1µν + G 2µν . By we mark the value up to the first order. The inverse of G µν is given by • Original background fields • Effective metric inverse • Theta function Θ µν (A.10)

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Using the explicit value of the initial metric the second term can be rewritten as 3) and therefore (B.4) So, the beta functions, defined by (3.7), are and in the light-cone coordinates they become

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The first two terms can be rewritten as Partially integrating, using (C.7), we obtain Finally, recalling (B.6) we obtain the dual beta functions