Courant bracket twisted both by a 2-form B and by a bi-vector θ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\theta $$\end{document}

We obtain the Courant bracket twisted simultaneously by a 2-form B and a bi-vector θ\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$\theta $$\end{document} by calculating the Poisson bracket algebra of the symmetry generator in the basis obtained acting with the relevant twisting matrix. It is the extension of the Courant bracket that contains well known Schouten–Nijenhuis and Koszul bracket, as well as some new star brackets. We give interpretation to the star brackets as projections on isotropic subspaces.


Introduction
The Courant bracket [1,2] represents the generalization of the Lie bracket on spaces of generalized vectors, understood as the direct sum of the elements of the tangent bundle and the elements of the cotangent bundle. It was obtained in the algebra of generalized currents firstly in [3]. Generalized currents are arbitrary functionals of the fields, parametrized by a pair of vector field and covector field on the target space. Although the Lie bracket satisfies the Jacobi identity, the Courant bracket does not.
In bosonic string theory, the Courant bracket is governing both local gauge and general coordinate transformations, invariant upon T-duality [4,5]. It is a special case of the more general C-bracket [6,7]. The C-bracket is obtained as the T-dual invariant bracket of the symmetry generator algebra, when the symmetry parameters depend both on the initial and T-dual coordinates. It reduces to the Courant bracket once when parameters depend solely on the coordinates from the initial theory.
It is possible to obtain the twisted Courant bracket, when the self T-dual generator algebra is considered in the basis  [8]. The Courant bracket is usually twisted by a 2-form B, giving rise to what is known as the twisted Courant bracket [9], and by a bi-vector θ , giving rise to the θ -twisted Courant bracket [10]. In [3,8,11,12], the former bracket was obtained in the generalized currents algebra, and it was shown to be related to the latter by self T-duality [13], when the Tdual of the B field is the bi-vector θ .
The B-twisted Courant bracket contains H flux, while the θ -twisted Courant bracket contains non-geometric Q and R fluxes. The fluxes are known to play a crucial role in the compactification of additional dimensions in string theory [14]. Non-geometric fluxes can be used to stabilize moduli. In this paper, we are interested in obtaining the Poisson bracket representation of the twisted Courant brackets that contain all fluxes from the generators algebra. Though it is possible to obtain various twists of the C-bracket as well [15], we do not deal with them in this paper.
The realization of all fluxes using the generalized geometry was already considered, see [16] for a comprehensive review. In [17], one considers the generalized tetrads originating from the generalized metric of the string Hamiltonian. As the Lie algebra of tetrads originating from the initial metric defines the geometric flux, it is suggested that all the other fluxes can be extracted from the Courant  In [18], one considers the standard Lie algebroid defined with the Lie bracket and the identity map as an anchor on the tangent bundle, as well as the Lie algebroid with the Koszul bracket and the bi-vector θ as an anchor on the cotangent bundle. The tetrad basis in these Lie algebroids is suitable for defining the geometric f and non-geometric Q fluxes. It was shown that by twisting both of these Lie algebroids by H -flux one can construct the Courant algebroid, which gives rise to all of the fluxes in the Courant bracket algebra.
Unlike previous approaches where generalized fluxes were defined using the Courant bracket algebra, in a current paper we obtain them in the Poisson bracket algebra of the symmetry generator.
Firstly, we consider the symmetry generator of local gauge and global coordinate transformations, defined as a standard inner product in the generalized tangent bundle of a double gauge parameter and a double canonical variable. The O(D, D) group transforms the double canonical variable into some other basis, in terms of which the symmetry generator can be expressed. We demonstrate how the Poisson bracket algebra of this generator can be used to obtain twist of the Courant bracket by any such transformation. We give a brief summary of how eB and eθ produce respectively the Btwisted and θ -twisted Courant bracket in the Poisson bracket algebra of generators [8].
Secondly, we consider the matrix eB used for twisting the Courant bracket simultaneously by a 2-form and a bi-vector. The argumentB is defined simply as a sum of the argumentŝ B andθ . UnlikeB orθ , the square ofB is not zero. The full Taylor series gives rise to the hyperbolic functions of the parameter depending on the contraction of the 2-form with the bi-vector α μ ν = 2κθ μρ B ρν . We represent the symmetry generator in the basis obtained acting with the twisting matrix eB on the double canonical variable. This generator is manifestly self T-dual and its algebra closes on the Courant bracket twisted by both B and θ .
Instead of computing the B − θ twisted Courant bracket directly, we introduce the change of basis in which we define some auxiliary generators, in order to simplify the calculations. This change of basis is also realized by the action of an element of the O(D, D) group. The structure constants appearing in the Poisson bracket algebra have exactly the same form as the generalized fluxes obtained in other papers [16][17][18]. The expressions for fluxes is given in terms of new auxiliary fieldsB andθ , both being the function of α μ .
The algebra of these new auxiliary generators closes on another bracket, that we callC-twisted Courant bracket. We obtain its full Poisson bracket representation, and express it in terms of generalized fluxes. We proceed with rewriting it in the coordinate free notation, where many terms are recognized as the well known brackets, such as the Koszul or Schouten-Nijenhuis bracket, but some new brackets, that we call star brackets, also appear. These star brackets as a domain take the direct sum of tangent and cotangent bundle, and as a result give the graph of the bi-vectorθ in the cotangent bundle, i.e. the sub-bundle for which the vector and 1-form components are related as ξ μ = κθ μν λ ν . We show that they can be defined in terms of the projections on isotropic subspaces acting on different twists of the Courant bracket.
Lastly, we return to the previous basis and obtain the full expression for the Courant bracket twisted by both B and θ . It has a similar form asC-twisted Courant bracket, but in this case the other brackets contained within it are also twisted. The Courant bracket twisted by both B and θ and the one twisted byC are directly related by a O(D, D) transformation represented with the block diagonal matrix.

The bosonic string essentials
The canonical Hamiltonian for closed bosonic string, moving in the D-dimensional space-time with background characterized by the metric field G μν and the antisymmetric Kalb-Ramond field B μν is given by [19,20] where π μ are canonical momenta conjugate to coordinates x μ , and is the effective metric. The Hamiltonian can be rewritten in the matrix notation where X M is a double canonical variable given by (2.4) and H M N is the so called generalized metric, given by with M, N ∈ {0, 1}. In the context of generalized geometry [21], the double canonical variable X M represents the generalized vector. The generalized vectors are 2D structures that combine both vector and 1-form components in a single entity.
The standard T-duality [22,23] laws for background fields have been obtained by Buscher [24] where (G −1 E ) μν is the inverse of the effective metric (2.2), and θ μν is the non-commutativity parameter, given by The T-duality can be realized without changing the phase space, which is called the self T-duality [13]. It has the same transformation rules for the background fields like Tduality (2.6), with additionally interchanging the coordinate σ -derivatives κ x μ with canonical momenta π μ κ x μ ∼ = π μ . (2.8) Since momenta and winding numbers correspond to σ integral of respectively π μ and κ x μ , we see that the self Tduality, just like the standard T-duality, swaps momenta and winding numbers.

Symmetry generator
We consider the symmetry generator that at the same time governs the general coordinate transformations, parametrized by ξ μ , and the local gauge transformations, parametrized by λ μ . The generator is given by [25] (2.9) It has been shown that the general coordinate transformations and the local gauge transformations are related by self Tduality [25], meaning that this generator is self T-dual. If one makes the following change of parameters λ μ → λ μ + ∂ μ ϕ, the generator (2.9) does not change (2.10) since the total derivative integral vanishes for the closed string. Therefore, the symmetry is reducible. Let us introduce the double gauge parameter M , as the generalized vector, given by where ξ μ represent the vector components, and λ μ represent the 1-form components. The space of generalized vectors is endowed with the natural inner product where i ξ is the interior product along the vector field ξ , and η M N is O(D, D) metric, given by Now it is possible to rewrite the generator (2.9) as (2.14) In [8], the Poisson bracket algebra of generator (2.9) was obtained in the form where the standard Poisson bracket relations between coordinates and canonical momenta were assumed where It is the generalization of the Lie bracket on spaces of generalized vectors.

O( D, D) group
Consider the orthogonal transformation O, i.e. the transformation that preserves the inner product (2.12) which is satisfied for the condition There is a solution for the above equation in the form O = e T , see Sec. 2.1 of [21], where  22) and note that the relation (2.15) can be written as and using (3.19) and (3.22) as where we expressed the right hand side in terms of some new bracket [ˆ 1 ,ˆ 2 ] C T . Moreover, using (3.19) and (3.22), the right hand side of (3.23) can be written as Using (3.24) and (3.25), one obtains This is a definition of a T -twisted Courant bracket. Throughout this paper, we use the notation where [, ] C is the Courant bracket, while when C has an additional index, it represents the twist of the Courant bracket by the indexed field, e.g.
[, ] C B is the Courant bracket twisted by B.
In a special case, when A = 0, θ = 0, the bracket (3.26) becomes the Courant bracket twisted by a 2-form B [9] where eB is the twisting matrix, given by This bracket has been obtained in the algebra of generalized currents [11,13].
In case of A = 0, B = 0, the bracket (3.26) becomes the Courant bracket twisted by a bi-vector θ where eθ is the twisting matrix, given by The B-twisted Courant bracket (3.27) and θ -twisted Courant bracket (3.29) are related by self T-duality [13]. It is easy to demonstrate that both eB and eθ satisfy the condition (3.20).
We can now deduce a simple algorithm for finding the Courant bracket twisted by an arbitrary O(D, D) transformation. One rewrites the double symmetry generator G(ξ, λ) in the basis obtained by the action of the matrix e T on the double coordinate (2.4). Then, the Poisson bracket algebra between these generators gives rise to the appropriate twist of the Courant bracket. In this paper, we apply this algorithm to obtain the Courant bracket twisted by both B and θ .

Twisting matrix
The transformations eB and eθ do not commute. That is why we define the transformations that simultaneously twists the Courant bracket by B and θ as eB, wherȇ The Courant bracket twisted at the same time both by a 2form B and by a bi-vector θ is given by The full expression for eB can be obtained from the well known Taylor series expansion of exponential function The square of the matrixB is easily obtained as well as its cubȇ The higher degree ofB are given by for even degrees, and for odd degrees by where we have marked Substituting (4.6) and (4.7) into (4.3), we obtain the twisting matrix Taking into the account the Taylor's expansion of hyperbolic functions the twisting matrix (4.9) can be rewritten as Its determinant is given by det(eB) = e T r(B) = 1, (4.12) and the straightforward calculations show that its inverse is given by (4.13) One easily obtains the relation therefore the transformation (4.

11) is indeed an element of O(D, D).
It is worth pointing out characteristics of the matrix α μ ν . It is easy to show that α for any analytical function f (α). Moreover, the well known hyperbolic identity cosh(x) 2 − sinh(x) 2 = 1 can also be expressed in terms of newly defined tensors Lastly, the self T-duality relates the matrix α to its transpose α ∼ = α T , due to (2.6). Consequently, we write the following self T-duality relations

Symmetry generator in an appropriate basis
The direct computation of the bracket (4.2) would be difficult, given the form of the matrix eB . Therefore, we use the indirect computation of the bracket, by computing the Poisson bracket algebra of the symmetry generator (2.9), rewritten in the appropriate basis. As elaborated at the end of the Chapter 3, this basis is obtained by the action of the matrix (4.11) on the double coordinate (2.4) Applying the transformation (4.11) to a double gauge parameter (2.11), we obtain new gauge parameters The symmetry generator (2.9) rewritten in a new basis G(Cξ + κSθλ, 2(BS)ξ + C T λ) ≡G(ξ,λ) is given by (5.23)

Auxiliary generator
Let us define a new auxiliary basis, so that both the matrices C and S are absorbed in some new fields, giving rise to the generator algebra that is much more readable. When the algebra in this basis is obtained, simple change of variables back to the initial ones will provide us with the bracket in need.
Multiplying the second equation of (5.19) with the matrix C −1 , we obtain where we have used (BS) νρ (C −1 ) ν μ = −(BSC −1 ) ρμ = (BSC −1 ) μρ , due to tensor BS being antisymmetric, and properties (4.15). We will mark the result as a new auxiliary current, given bẙ whereB is an auxiliary B-field, given bẙ On the other hand, multiplying the first equation of (5.19) with the matrix C, we obtain Substituting (4.16) in the previous equation, and keeping in mind that C, S and θ commute (4.15), we obtain Using (5.25), the results are marked as a new auxiliary current whereθ is given bẙ There is no explicit dependence on either C nor S in redefined auxiliary currents, rather only on canonical variables and new background fields. From (5.29), it is easy to express the coordinate σ -derivative in the basis of new auxiliary currents The first equation of (5. 19) could have been multiplied with C, instead of C −1 , given that the latter would also produce a current that would not explicitly depend on C. However, the expression for coordinate σ -derivative κ x μ would explicitly depend on C 2 in that case, while with our choice of basis it does not (5.31).
Substituting (5.24) and (5.28) in the expression for the generator (5.22), we obtain from which it is easily seen that the generator (5.22) is equal to an auxiliary generator provided that and Once that the algebra of (5.33) is known, the algebra of generator (5.22) can be easily obtained using (5.34).
The change of basis to the one suitable for the auxiliary generator (5.33) corresponds to the transformation that can be rewritten as where theC-twisted Courant bracket is defined by In the next chapter, we will obtain this bracket by direct computation of the generators Poisson bracket algebra. Lastly, let us briefly comment on reducibility conditions for theC-twisted Courant bracket. Since we are working with the closed strings, the total derivatives vanishes when integrated out over the worldsheet. Using (5.31), we obtain These are reducibility conditions (2.10) in the basis spanned byk μ andι μ .

Courant bracket twisted byC from the generator algebra
In order to obtain the Poisson bracket algebra for the generator (5.33), let us firstly calculate the algebra of basis vectors, using the standard Poisson bracket relations (2.16). The auxiliary currentsι μ algebra is whereB μνρ is the generalized H-flux, given bẙ andF ρ μν is the generalized f-flux, given bẙ 3) The algebra of currentsk μ is given by The terms in (6.4) containing bothθ andB are the consequence of non-commutativity of auxiliary currentsι μ . The remaining algebra of currentsk μ andι μ can be as easily obtained The basic algebra relations can be summarized in a single algebra relation where the structure constants contain all generalized fluxes The form of the generalized fluxes is the same as the ones already obtained using the tetrad formalism [16][17][18]. In our approach, the generalized fluxes are obtained in the Poisson bracket algebra, only from the fact that the generalized canonical variable X M is transformed with an element of the O(D, D) group that twists the Courant bracket both by B and θ at the same time. Consequentially, the fluxes obtained in this paper are functions of some new effective fields,B μν (5.26) andθ μν (5.30).
We now proceed to obtain the full bracket. Let us rewrite the generator (5.33) algebra 10) The first term of (6.10) is obtained, using (6.1) The second term is obtained, using (6.4) The remaining terms are antisymmetric with respect to 1 ↔ 2, σ ↔σ interchange. Therefore, it is sufficient to calculate only the first term in the last line of (6.10) In order to transform the anomalous part, we note that and Applying (6.14) and (6.15) to the last row of (6.13), we obtain where (5.31) was used, as well as antisymmetry ofθ . Substituting (6.16) to (6.13), we obtain Substituting (6.11), (6.12) and (6.17) into (6.10), we write the full algebra of generator in the form G (ξ 1 ,λ 1 ),G(ξ 2 ,λ 2 ) = −G(ξ,λ), and It is possible to rewrite the previous two equations, if we note the relations between the generalized fluxes R μνρ =R μνρ +θ μσθ ντF ρ σ τ ,Q νρ μ =Q νρ μ +θ νσF ρ μσ . (6.21) Now we have and where the partial integration was used in the equation (6.22). The relation (6.18) defines theC-twisted Courant bracket (6.24) that gives the same bracket as (5.41). Both (6.19)-(6.20) and (6.22)-(6.23) are the products ofC-twisted Courant bracket. The former shows explicitly how the gauge parameters depend on the generalized fluxes. In the latter, similarities between the expressions for two parameters is easier to see.

Special cases and relations to other brackets
Even though the non-commutativity parameter θ and the Kalb Ramond field B are not mutually independent, while obtaining the bracket (6.24) the relation between these fields (2.7) was not used. Therefore, the results stand even if a bi-vector and a 2-form used for twisting are mutually independent. This will turn out to be convenient to analyze the origin of terms appearing in the Courant bracket twisted bẙ C.
Primarily, consider the case of zero bi-vector θ μν = 0 with the 2-form B μν arbitrary. Consequently, the parameter α (4.8) is zero, while the hyperbolic functions C and S are identity matrices. Therefore, the auxiliary fields (5.26)  and where B μνρ is the Kalb-Ramond field strength, given by The equations (6.26) and (6.27) define exactly the B-twisted Courant bracket (3.27) [9]. Secondarily, consider the case of zero 2-form B μν = 0 and the bi-vector θ μν arbitrary. Similarly, α = 0 and C and S are identity matrices. The auxiliary fieldsB μν andθ μν are given bẙ B μν → 0θ μν → θ μν . (6.29) The twisting matrix eB becomes the matrix of θ -transformations eθ (3.30). The gauge parameters (6.19) and (6.20) are respec-tively given bẙ and where by Q νρ μ and R μνρ we have marked the non-geometric fluxes, given by The bracket defined by these relations is θ -twisted Courant bracket (3.29) [8] and it features the non-geometric fluxes only. Let us comment on terms in the obtained expressions for gauge parameters (6.22) and (6.23). The first line of (6.22) appears in the Courant bracket and in all brackets that can be obtained from its twisting by either a 2-form or a bi-vector. The next two lines correspond to the terms appearing in the θ -twisted Courant bracket (6.30). The other terms do not appear in either B-or θ -twisted Courant bracket.
Similarly, the first line of (6.20) appears in the Courant bracket (2.18) and in all other brackets obtained from its twisting, while the terms in the second line appear exclusively in the θ twisted Courant bracket (6.27). The first term in the last line appear in the B-twisted Courant bracket (6.31), while the rest are some new terms. We see that all the terms that do not appear in neither of two brackets are the terms containing F flux.

Coordinate free notation
In order to obtain the formulation of theC-twisted Courant bracket in the coordinate free notation, independent of the local coordinate system that is used on the manifold, let us firstly provide definitions for a couple of well know brackets and derivatives.

Star brackets
The expressions for gauge parameters (6.36) and (6.37) produce some well known bracket, such as Lie bracket and Koszul bracket. The remaining terms can be combined so that they are expressed by some new brackets, acting on pairs of generalized vectors. It turns out that these brackets produce a generalized vector, where the vector partξ μ and the 1-form partλ μ are related byξ μ = κθ μνλ ν , effectively resulting in the graphs in the generalized cotangent bundle T M of the bi-vectorθ, i.e. ξ = κθ(., λ). The star brackets can be interpreted in terms of projections on isotropic subspaces.

θ -star bracket
Let us firstly consider the second line of (6.22) and the first line of (6.23). When combined, they define a bracket acting on a pair of generalized vectors and from which one easily reads the relation In a coordinate free notation, this bracket can be written as The remaining terms contain geometricH andF fluxes. Note that they are the only terms that depend on the new effective Kalb-Ramond fieldB. Firstly, we mark the last line of (6.23) as Secondly, using the definition ofF (6.3) and the fact thatθ is antisymmetric, the last line of (6.22) can be rewritten as Now relations (7.6) and (7.7) define the Bθ -star bracket by [˚ 1 ,˚ 2 ] * Bθ =˚ * ⇔ [(ξ 1 ,λ 1 ), (ξ 2 ,λ 2 )] * Bθ = (ξ * ,λ * ), (7.8) We can write the full bracket (6.24) as

Isotropic subspaces
In order to give an interpretation to newly obtained starred brackets, it is convenient to consider isotropic subspaces. A subspace L is isotropic if the inner product (2.12) of any two generalized vectors from that sub-bundle is zero From (2.12), one easily finds that ξ μ i = κ θ μν λ iν . (i = 1, 2) θ μν = −θ νμ , (7.11) for any bi-vector θ , and (7.12) for any 2-form B satisfy the condition (7.10). Furthermore, it is straightforward to introduce projections on these isotropic subspaces by I θ ( M ) = I θ (ξ μ , λ μ ) = (κ θ μν λ ν , λ μ ), (7.13) and Now it is easy to give an interpretation to star brackets. The θ -star bracket (7.1) can be defined as the projection of the Courant bracket (3.29) on the isotropic subspace (7.13) Similarly, note that all the terms in (6.37) that do not appear in the θ -twisted Courant bracket, contribute exactly to the Bθ -star bracket. From that, it is easy to obtain the definition of the Bθ -star bracket (7.8)

Courant bracket twisted by B and θ
Now it is possible to write down the expression for the Courant bracket twisted by B and θ (4.2), using the expression forC-twisted Courant bracket where A is defined in (5.36). Substituting (8.1) into (6.36), we obtain +C −1 ∧ 2 κθH (λ 2 C −1 , ., Cξ 1 ) and similarly, substituting (8.1) into (6.37), we obtain where C μ ν = cosh √ α μ ν and˘ = (ξ,λ) (5.21). This is somewhat a cumbersome expression, making it difficult to work with. To simplify it, with the accordance of our convention, we define the twisted Lie bracket by as well as the twisted Schouten-Nijenhuis bracket and twisted Koszul bracket where the transpose of the matrix is necessary because the Koszul bracket acts on 1-forms. Now, the first three terms of (8.2) can be written as wherȇ The second line of (8.2) and the first line of (8.3) originating fromθ star bracket (7.1) can be easily combined into The terms originating fromBθ star bracket (7.8) are combined into wherȇ The expressions for the Courant bracket twisted by both B and θ can be written in a form When the Courant bracket is twisted by both B and θ , it results in a bracket similar toC-twisted Courant bracket, where Lie brackets, Schouten Nijenhuis bracket and Koszul bracket are all twisted as well.

Conclusion
We examined various twists of the Courant bracket, that appear in the Poisson bracket algebra of symmetry generators written in a suitable basis, obtained acting on the double canonical variable (2.4) by the appropriate elements of O(D, D) group. In this paper, we considered the transformations that twists the Courant bracket simultaneously by a 2-form B and a bi-vector θ . When these fields are mutually T-dual, the generator obtained by this transformation is invariant upon self T-duality. We obtained the matrix elements of this transformation, that we denoted eB (4.11), expressed in terms of the hyperbolic functions of a parameter α (4.8). In order to avoid working with such a complicated expression, we considered another O(D, D) transformation A (5.36) and introduced a new generator, written in a basis of auxiliary currentsι μ andk μ . The Poisson bracket algebra of a new generator was obtained and it gave rise to theC-twisted Courant bracket, which contains all of the fluxes.
The generalized fluxes were obtained using different methods [10][11][12][16][17][18]. In our approach, we started by an O(D, D) transformation that twists the Courant bracket simultaneously by a 2-form B and bi-vector θ , making it manifestly self T-dual. We obtained the expressions for all fluxes, written in terms of the effective fields The fluxes, as a function of these effective fields, appear naturally in the Poisson bracket algebra of such generators.
Similar bracket was obtained in the algebra of generalized currents in [11,12] and is sometimes referred to as the Roytenberg bracket [10]. In that approach, phase space has been changed, so that the momentum algebra gives rise to the H -flux, after which the generalized currents were defined in terms of the open string fields. The bracket obtained this way corresponds to the Courant bracket that was firstly twisted by B field, and then by a bi-vector θ . The matrix of that twist is given by In our approach, we obtained the transformations that twists the Courant bracket at the same time by B and θ , resulting in å C-twisted Courant bracket. As a consequence, theC-twisted Courant bracket is defined in terms of auxiliary fieldsB (5.26) andθ (5.30), that are themselves function of α. This is not the case in [11,12]. The Roytenberg bracket calculated therein can be also obtained following our approach by twisting with the matrix demanding that the background fields are infinitesimal B ∼ , θ ∼ and keeping the terms up to 2 . With these conditions, e C (9.3) becomes exactly e R (9.2), and the bracket becomes the Roytenberg bracket.
Analyzing theC-twisted Courant bracket, we recognized that certain terms can be seen as new brackets on the space of generalized vectors, that we named star brackets. We demonstrated that they are closely related to projections on isotropic spaces. It is well established that the Courant bracket does not satisfy the Jacobi identity in general case. The sub-bundles on which the Jacobi identity is satisfied are known as Dirac structures, which as a necessary condition need to be subsets of isotropic spaces. Therefore, the star brackets might provide future insights into integrability conditions for the C-twisted Courant bracket [28].
In the end, we obtained the Courant bracket twisted at the same time by B and θ by considering the generator in the basis spanned byι andk, equivalent to undoing A transformation, used to simplify calculations. With the introduction of new fieldsB μν andθ μν , this bracket has a similar form asC-twisted Courant bracket, whereby the Lie, Schouten-Nijenhuis and Koszul brackets became their twisted counterparts.
It has already been established that B-twisted and θtwisted Courant brackets appear in the generator algebra defined in bases related by self T-duality [13]. When the Courant bracket is twisted by both B and θ , it is self T-dual, and as such, represent the self T-dual extension of the Lie bracket that includes all fluxes. It has been already shown [8] how the Hamiltonian can be obtained acting with Btransformations on diagonal generalized metric. The same method could be replicated with the twisting matrix eB, that would give rise to a different Hamiltonian, whose further analysis can provide interesting insights in the role that the Courant bracket twisted by both B and θ plays in understanding T-duality.

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