SciELO - Scientific Electronic Library Online

vol.40 número4Aspects of nonmetricity in gravity theories2d Gravity with torsion, oriented matroids and 2+2 dimensions índice de autoresíndice de materiabúsqueda de artículos
Home Pagelista alfabética de revistas  

Servicios Personalizados




Links relacionados


Brazilian Journal of Physics

versión impresa ISSN 0103-9733

Braz. J. Phys. vol.40 no.4 São Paulo dic. 2010 

Conformal field theory with two kinds of bosonic fields and two linear dilatons



Davoud Kamani*

Faculty of Physics, Amirkabir University of Technology (Tehran Polytechnic) P.O.Box: 15875-4413, Tehran, Iran




We consider a two-dimensional conformal field theory which contains two kinds of the bosonic degrees of freedom. Two linear dilaton fields enable us to study a more general case. Various properties of the model such as OPEs, central charge, conformal properties of the fields and associated algebras will be studied.

Keywords: String; Linear Dilaton CFT; OPE.




Among the various conformal field theories (CFTs) the linear dilaton CFT has some interesting applications in the string theory, e.g. see [1-6]. In this CFT, modification of the energy-momentum tensor was anticipated by a linear dilaton field. This CFT significantly changes the behavior of the worldsheet theory. In addition, this CFT is a consistent way for reducing the spacetime dimension without compactification. The linear dilaton CFT also appears as an ingredient in many string backgrounds, critical and non-critical. According to its importance we proceed to develop it.

In this paper we consider an action which is generalization of the bosonic part of the = 2 superstring theory. In addition, we introduce two linear dilaton fields to build our model. Thus, we study a conformally invariant field theory in two flat dimensions. Anticipating to the string theory, we refer to these two dimensions as the string worldsheet. Various OPEs of the model will be calculated. Due to the dilaton fields, some of these OPEs, and also conformal transformations of the worldsheet fields Xµ(σ, τ) and Yµ(σ, τ) have deviations from the standard forms. Presence of some parameters in the central charge enables us to receive a desirable dimension for the spacetime. The algebra of the oscillators reveals that the oscillators of X-fields do not commute with that of Y-fields.

This paper is organized as follows. In section 2, we shall introduce the action of the model and the linear dilatonic energy-momentum tensor associated to it. In section 3, various OPEs of the model will be studied. In section 4, conformal transformations of the worldsheet fields will be obtained. In section 5, various quantities will be expressed in terms of the oscillators, and two algebras for the model will be obtained. Section 6 is devoted for the conclusions.



We begin with the action of the scalar fields Xµ (z, ) and Yµ (z, ) in two dimensions

where µ {0,1,...,D-1} and β and λ are constants, i.e. independent of z and . For the spacetime we consider the flat Minkowski metric ηµν = diag(-1,1,...,1) . The special case β = 1 and λ = 0 indicates the bosonic part of the = 2 super-conformal field theory. Thus, we say the set {Xµ } describes the spacetime coordinates. In other words, Xµ (σ, τ) is regarded as the embedding of the worldsheet in the spacetime. However, Yµ (σ, τ) enters essentially in the same way. So the set {Yµ (σ, τ)} does not describe additional dimensions. The conformal invariance of this action, i.e. symmetry under the conformal transformations z z'(z) and '(), leads to the zero conformal weights for the fields Xµ and Yµ.

The equations of motion, extracted from the action (1), are

We assume that the determinant of the coefficients of these equations to be nonzero i.e.,

Therefore, we obtain

These imply zXµ and zYµ are functions of z, and Xµ and Yµ are functions of .

The corresponding energy-momentum tensor has the components

where : : denotes normal ordering.

It is possible to construct a more general CFT with the same action (1), but with different energy-momentum tensor

where sum over i and j is assumed with i, j {1,2}. We define

The vectors Vm and Um are fixed in the spacetime. For each pair of these vectors we have a CFT. The extra terms in (6) are total derivatives. Thus, we shall see that they do not affect the status of T(z) and () as generators of conformal transformations. The field Φ = Vµ Xµ in (6) is linear dilaton. In the same way Φ' = Uµ Yµ is a linear field in the Y-space. In fact, by introducing the worldsheet fields {Yµ (σ, τ)} and defining the energy-momentum tensor (6), we have generalized the linear dilaton CFT. The case β = 1 and λ = 0 decomposes the model to two copies of the linear dilaton CFT.



3.1. The OPEs XX, XY and YY

We use the path integral formalism to derive operator equations. Since the path integral of a total derivative is zero, we have the equation

The point (w, ) might be coincident with (z, ), but the insertion " ... " is arbitrary, which is away from (z ,) and (w, ). Arbitraryness of the insertion implies

as an operator equation. In the same way, the equation

gives the operator equation

In the equation (10) change Xµ to Yµ, we obtain

Similarly, in the first line of (8) replacing Xµ to Yµ

The equations (9), (11), (12) and (13) give the following equations

That is, the equations of motion (4) hold except at the coincident point (z, ) = (w, ). Define the matrix Qij as in the following

Thus, the equations (14) can be written in the compact form

According to this, we have the normal ordered equation

where z ln|z — w|2 = 2πδ(2)(z — w, ) has been used. The equation (16) and (17) indicate the equation of motion

3.2 The TT OPE

Let be any functional of {Xµ} and {Yµ}. Thus, the generalization of (17) is defined by

The OPE for any pair of the operators and is given by

where the functional derivatives act only on the fields or , respectively. For = Xµi (z , ) and = Xnj(w,) this reduces to the equation (17), as expected.

Using the equation (20), we obtain

Now the Taylor expansion of z Xµi(z) around z = w changes this equation to

where the non-singular terms have been omitted. For calculating the TT OPE we also need the following OPEs

Adding all these together we obtain the TT OPE as in the following

The OPE also has a similar form in terms of , and .

The central charges are given by

Vanishing conformal anomaly relates the parameters of the model. That is, string actually can move in a wide range of the dimensions. However, by adjusting the variables β, λ, Vµ and Uµ, we can obtain desirable dimension for the spacetime. The case Vµ = Uµ = 0 gives the central charges c = = 2D, i.e., D for {Xµ} and D for {Yµ}. If β = 1 and λ = 0, the action (1) reduces to two copies of the free string action, and hence the energy-momentum tensor (6) is modified to two copies of the energy-momentum tensor of the linear dilaton CFT. In this case the central charge also reduces to two copies of the central charge of the linear dilaton CFT

Since there is ΛQ = I2×2, the TT OPE (26), and similarly the OPE take the standard forms

According to the central charge terms, T and are not conformal tensors. Apart from these terms, (29) is the statement that T(z) and () are conformal fields of the weights (2,0) and (0,2), respectively.

3.3 The OPEs TX, TY, X and Y

The OPE TXkµ is

Thus, for k = 1 and k = 2 we obtain

In the same way we have

The U-terms and V-terms imply that Xµ and Yµ are not conformal tensor operators. Putting away these terms (the square singular terms) of the above OPEs leads to the conditions

Since we assumed βλ2 0, we obtain Vµ = Uµ = 0. Therefore, (31) and (32) reduce to the OPEs T'X, T'Y, 'X and 'Y. That is, with T' and ' the fields Xµ and Yµ are conformal tensors, as expected. However, we shall not consider the case (33).



The infinitesimal conformal transformations z z' = z+εg(z) and ' = '+εg(z)* imply the currents

For any holomorphic function g(z) these are conserved. These currents lead to the Ward identity

where "Res" and "" are coefficients of (z–w)-1 and ()-1, respectively. From the OPEs (31) and (32) and the Ward identity (35) we obtain the conformal transformations

Due to the inhomogeneous parts, originated from Vµ, Uµ, β and λ, the fields Xµ and Yµ do not transform as conformal tensor. These parts also indicate that these transformations are not infinitesimal coordinate transformations δz = εg(z) and δz = εg(z)*.



Now we express some quantities of the model in terms of the oscillators of Xµ and Yµ. The OPEs (31) and (32) give

Thus, the conformal weights of zXµ (z) and zYµ (z) are

According to these conformal weights, we obtain the Laurent expansions

Single-valuedness of Xµ and Yµ implies that

where pµi is the linear momentum. Now integration of the expansions (41) gives the closed string solution

Reality of Xµi implies that ᵆ(i)m = αµ(i)(-m) and µ†(i)m = µ(i)(-m).

The expansions (41) also lead to

where C in the z-plane and in the -plane are counterclockwise. Therefore, by using the OPEs zXµi(z)wXνj(w) and Xµi()Xνj() we obtain

For λ 0 we observe that the oscillators of Xµ do not commute with the oscillators of Yµ.

In terms of the oscillators the nonzero elements of the energy-momentum tensor find the forms

The Virasoro operators are

In terms of the oscillators they take the forms

Using the standard methods one can show that the normal ordering constant for all Lm and m is zero. According to the equations (45), or the standard form of the OPEs TT and , i.e. the equations (29), the Virasoro algebra also has the standard form

The Hamiltonian of the system is given by

Thus, the equations (27) and (48) express this Hamiltonian in terms of the oscillators and the parameters of the model

where the symmetry of ηµν and Λij were introduced.

For the open string there are

and hence the solution is

The corresponding energy-momentum tensor and Virasoro operators are given by the first equations of (46) and (48). Thus, the associated Virasoro algebra also is described by the first equation of (49).

Note that we imposed the boundary conditions of the closed string and open string on Yµ (σ, τ). However, Yµ (σ, τ) may be neither closed nor open. Assuming closeness or openness for Yµ (σ, τ), the worldsheet fields (Xµ (σ, τ) , Yµ (σ, τ)) find four configurations: (closed , closed), (open , open), (open , closed) and (closed , open). We considered the first and the second cases. The third and the fourth cases also can be investigated in the same way.



We studied a CFT model with two kinds of the bosonic degrees of freedom Xµ and Yµ, which interact kinetically with each other. For each kind of these fields we introduced a linear dilaton field.

Using the path integral formalism, we obtained the OPEs XX, XY and YY. These OPEs enabled us to introduce a general definition for the OPEs. We observed that the TT and OPEs of the model have the standard forms. Due to the vectors Vµ and Uµ, which define the dilatons, the OPEs TX, TY, X and Y have deviations from the standard forms of them. The central charge of the model depends on the spacetime dimension, the parameters of the theory and the vectors Vµ and Uµ. A vanishing conformal anomaly and hence a desirable dimension for the spacetime can be achieved by tuning these variables.

Putting away the interacting terms of the action, the model split into two copies of the linear dilaton CFT. The splitting also occurs for the energy-momentum tensor and hence for the central charge.

Using the conserved currents, associated to the conformal symmetry, the conformal transformations of the fields Xµ and Yµ have been extracted. Therefore, the vectors Vm and Um and also the parameters of the model indicate that Xµ and Yµ are not conformal tensors. That is, these transformations are not pure coordinate transformations.

According to the mode expansions of Xµ and Yµ, we obtained the oscillator-algebra of the model. Due to the nonzero coupling constant λ the oscillators of Xµ do not commute with the oscillators of Yµ. We expressed the energy-momentum tensor and the Virasoro operators in terms of the oscillators. We observed that the Virasoro operators also form the standard algebra.


[1] T. Takayanagi, JHEP 0412 (2004) 071, hep-th/0411019; JHEP 0509 (2005) 001, hep-th/0507065.         [ Links ]

[2] S. Nakamura and V. Niarchos, JHEP 10 (2005) 025.         [ Links ]

[3] O. Bergman and S. Hirano, Nucl. Phys. 744 (2006) 136.         [ Links ]

[4] Y. Hikida, K. Hosomichi and Y. Sugawara, Nucl. Phys. B589 (2000) 134.         [ Links ]

[5] P.M. Ho, S.Y. Darren Shih, JHEP 0801 (2008) 054, arXiv:0711.2792.         [ Links ]

[6] M. Li, Phys. Rev. D54 (1996) 1644, hep-th/9512042.         [ Links ]



(Received on 26 June, 2009)

Creative Commons License Todo el contenido de esta revista, excepto dónde está identificado, está bajo una Licencia Creative Commons