String field representation of the Virasoro algebra

We construct a representation of the zero central charge Virasoro algebra using string fields in Witten's open bosonic string field theory. This construction is used to explore extensions of the KBc algebra and find novel algebraic solutions of open string field theory.


Introduction
Our theory of interest is Witten's open bosonic string field theory [1]. In particular, we focus on the research inspired by [2], where this theory was used to prove that the energy of the tachyon vacuum is minus the energy of the D-25 brane. There has been a good deal of progress made towards simplifying the original tachyon vacuum solution [3,4]. This simple solution is expressed in a language which makes use of an algebra of string fields called the KBc algebra. Despite the advantages of this approach, there are various problems that can arise when using the KBc algebra to construct solutions other than the tachyon vacuum [5,6,7,8]. Our attitude in this work is that these problems arise because the KBc algebra is not large enough to properly describe all solutions of open string field theory.
If one tries to construct an algebra of string fields in an arbitrary way, the star products between the elements will be too difficult to manage. Therefore, in order to extend the KBc algebra in a meaningful way, we must ask the question: Under what conditions can one straightforwardly construct an algebra of string fields with manageable star products? In the rest of this section we introduce one such family of states with simple star product structure.
Consider the operator modes φ n corresponding to a primary conformal field φ(z) of weight h. These modes may be written as where the contour of integration is along the complex unit circle unless otherwise specified. If we make a conformal transformationz = f (z), then the transformed modesφ n are given byφ It is convenient to introduceṽ n (z) = ∂f (z) −h+1 [f (z)] n+h−1 , so we havẽ The modesφ n can be decomposed into their left and right components, respectively given byφ where L denotes integration along the Re(z) > 0 half of the complex unit circle and R denotes integration along the Re(z) < 0 half of the complex unit circle 1 . Therefore, the sum of the left and right components corresponds to integration along the entire complex unit circle, namely,φ L n +φ R n =φ n . The left and right components of operators are interesting objects in string field theory because of their convenient properties with respect to the star product. For any string fields A and B, we have where in the last line |A| and |φ| refer to the ghost number of A and φ, respectively. We now focus our attention to the left componentsφ L n . Let us define the string fields where |I is the identity of the star product. Using (5), we can compute the star commutator We note that in the above manipulation |Φ L n | = |φ L n |, since |I has ghost number zero. Also, it will be assumed throughout that commutators are graded by ghost number. The result (7) shows us that if we create an algebra of string fields with elements Φ L n , then the star commutators can be entirely determined by evaluating the ordinary commutators [φ L m ,φ L n ]. We now provide an explanation of the conditions under which (7) can be written in terms of a closed algebra of string fields.
Suppose that φ(z) belongs to a family of primary conformal fields indexed by a set J, φ(z) ∈ {φ α (z)} α∈J , such that where the f α mn are constants and the modes φ α n correspond to φ α (z). An important observation of this work is that there sometimes exists a conformal framez in which φ n andφ L n satisfy the same algebra, meaning that where the constants f α mn are the same in both cases. 2 In this situation, it is straightforward to see that We refer to the algebra generated by (10) as the string field representation of the algebra (8) with structure constants f α mn . This result answers the question posed at the beginning of this discussion. In particular, the condition (9) allows one to straightforwardly construct an algebra of string fields with manageable star products. 3 The main observation of this work is that we have precisely the condition (9) for the matter plus ghost Virasoro modes L n and the conformal framez = 2 π arctan z. The modes L n satisfy the zero central charge Virasoro algebra, which we now refer to simply as the Virasoro algebra. If we letL n = L n and define the string fields We call the algebra generated by (11) the string field representation of the Virasoro algebra. Naively, one would expect this discussion to be exactly the same for the right components. It is true that the modes L R n satisfy the Virasoro algebra, however, there is one interesting subtlety. Define the string fields L * n = L R n |I . Using the rule Recall that the BPZ dual of L n is given by L * n = (−1) n L −n . Therefore, the BPZ dual algebra is [L * m , L * n ] = −(m − n)L * m+n . We see from this observation that the algebra generated by (12) is actually the string field representation of the BPZ dual algebra.
This paper is outlined as follows. In section 2, we prove the claim that L n together with the conformal framez = 2 π arctan z satisfy the condition (9). We also discuss complications which arise if one considers correlation functions with operator insertions at the open string midpoint. In section 3, we discuss various options for extending the KBc algebra. In section 4, we use our results to find novel algebraic solutions of open string field theory. We conclude with a brief summary of our results and comment on opportunities for future exploration.

Left and right components of L n
Since we already know that [L m , L n ] = (m − n)L m+n , the main goal of this section is to show that [L L m , L L n ] = (m − n)L L m+n . The first step towards showing these com-mutation relations is to explicitly express the operator modes L n as For the sake of brevity, we define An important property of the vector fields v n (z) is that A quick but a bit formal argument for where we have introduced the 'holomorphic step function' satisfying θ(Re(z)) = 1 for Re(z) > 0 and θ(Re(z)) = 0 for Re(z) < 0. Let us define L v = dz 2πi v(z)T (z). Formally, or under suitable conditions, for any two such operators [L v , L w ] = −L [v,w] , where [v, w] = v∂w − w∂v denotes the Lie bracket. Applying this formula for two vector fields of the form v n (z)θ(Re(z)) one quickly establishes and the formal properties of the holomorphic step function θ(Re(z)) 2 = θ(Re(z)) and ∂ z θ(Re(z)) = 0, where especially the latter one may seem dubious. Because of central importance of the equation (18) to this work, let us present a more rigorous derivation. To proceed we follow the standard contour argument with modifications due to the step functions which restrict both contours to semicircles Figure 1: Contour manipulation involved in proving (18). The blue z-contour is deformed from C R 1+ε into C R 1−ε leaving behind small circle around the singularity at w, and integration along two open vertical segments of length 2ε. The variable w is integrated along the unit red semicircle. as in Figure 1. By picking sufficiently small ε > 0, the commutator can be expressed as In analogy to the standard argument we can deform the z-variable contour C R 1+ε into the C R 1−ε contour so that they cancel each other. What remains is a sum of two terms I 1 + I 2 The first term I 1 is given by a small contour C w around the point w. Only the singular part of the zero-central-charge OPE contributes. The resulting contribution takes the form where in the second line we used integration by parts. The first term already accounts for our desired commutation relation (18) thanks to (19). The last two terms are a contribution from the ends of the contour. They vanish since v n (±i) = 0, but this computation also hints at possible problems. Inserting the term I 1 inside a correlator with generic mid-point insertions at ±i, the explicit appearance of T (±i) on the right hand side of (24) would lead to divergences and the final result would depend on the precise manner the various limits are taken. In this work we allow the probing operator to approach the midpoint at the very end, so that the midpoint contributions in (24) are effectively absent. The second term I 2 is naively not contributing either, since the integration region is of vanishing size as ε is taken to zero. One must exercise a caution however, since the integrand of the double integral (22) is divergent in the region z ∼ w ∼ ±i where its leading singularity is given by Here we parameterized z = ±i + it and w = ±i + u. Standard power-counting argument-assuming regular T (u)-shows however that the singularity is integrable, and hence the contribution from a vanishing size region is indeed vanishing. The easiest way to see this is by passing to radial coordinates in the t-u plane. On the other hand, had we evaluated I 2 inside a correlator with midpoint insertions, we would have to replace T (u) by e.g. 1/u 2 in case of a primary field, and I 2 would have been divergent, or at least prescription dependent. Let us close this section by noting that similarly to (16), we have where θ(Re(−z)) corresponds to integration along the Re(z) < 0 half of the complex unit circle. We find the expected result One may also consider commutators involving both left and right components. Using a similar analysis, we obtain 4 [L L m , L R n ] = 0.

Extensions of the KBc algebra
We first recall the most important results of sections 1 and 2. We have shown that the strings fields L n = L L n |I form a representation of the Virasoro algebra We have also seen that the string fields L * n = L R n |I form a representation of the BPZ dual algebra At this point we restrict our discussion for convenience to the Virasoro algebra rather than its dual. However, similar remarks will hold if one wishes to formulate a theory using the BPZ dual algebra. The string fields of the KBc algebra are defined in our language as where as before the tilde refers to the operator expressed in thez = 2 π arctan z conformal frame. Given our previous observations, it is clear that we may define an algebra of anticommuting string fields analogous to B, given by where ∂c =∂c 1 2 |I . We are now prepared to begin our discussion of extending the KBc algebra. The most straightforward extension is to include all of the string fields L n and B n . This algebra satisfies The commutator [L n , c] is a bit trickier to evaluate. We begin by computing Using the rule (c 1 2 |I ) ⋆ (L n |I ) =c 1 2 L n |I , we see that By computing the commutator (36), we find and hence Qc = (2) n+1 c L n c.
Notice that by defining C n = (2) n+1 c, we have The above relationships will be convenient when we use these results to write down solutions of open string field theory. Another possibility is to consider a finite extension of the KBc algebra. In fact, a finite extension is often computationally easier to understand. The infinite extension was introduced first in order to develop all of the techniques necessary to deal with extended KBc algebras. The Virasoro algebra has two non-trivial finite subalgebras. The elements L −1 and L 0 form what is called aff(1), while L −1 , L 0 , and L 1 form the familiar SL(2, R) algebra. By adding the B counterparts to either aff(1) or SL(2, R), one can create a finite extension of the KBc algebra. However, it should be noted that one is not strictly limited to these cases. For the generating string fields one could instead choose various linear combinations of the elements in aff (1) or SL(2, R). In fact, one of the early motivations for this work was the discovery of one of the aff(1) linear combinations. Consider the string field The string field L has the interesting property that where L − = 1 2 (L 0 − L * 0 ) is the familiar derivation of the star algebra. Therefore, adding L to the KBc algebra is effectively turning an exterior derivative into an interior derivative.
The SL(2, R) extension also has a nice physical interpretation. It is well-known that the string field K acts as a generator of translations when acting on the string field c, a fact which is expressed by the commutation relation [K, c] = ∂c. It turns out that the SL(2, R) extension effectively adds the generators of dilation and special conformal transformation to the KBc algebra. To see this, let us use the convention that the generator G n associated with L n is defined implicitly by [L n , c] = iG n c. Then we see from (39) that G n = −i − (n + 1)z n +z n+1∂ , where we letz → 1 2 . Notice that the generators G −1 , G 0 , and G 1 form a representation of the holomorphic component of the global conformal algebra in two dimensions.

Application to algebraic solutions
The goal of this section is to show that we can use the extensions described in section 3 to construct new analytic solutions to the open string field theory equation of motion QΨ + Ψ ⋆ Ψ = 0. We begin by reviewing important techniques for constructing solutions with the KBc algebra. The modern method of constructing solutions is to start with the pure gauge ansatz U = 1 − F BcF , where F = F (K) is an appropriate function [14] of the string field K. The corresponding solution Ψ is given by Ψ = UQU −1 . In order to find U −1 , we compute This result for U −1 leads to the solution which is the familiar Okawa ansatz discovered in [3].
In the spirit of section 3, we first show how this solution nicely generalizes to the infinite extension of KBc, which includes all of the string fields L n , B n , and C n . We start with the pure gauge ansatz for a fixed choice of n. The relationships (34) and (39) tell us that for each fixed value of n, the L n , B n , C n algebra behaves almost identically to the original KBc algebra. Therefore, we find that the pure gauge ansatz U n leads to the solution The computation and classification of all possible solutions using different representations of the KBc algebra is certainly a project in itself, and therefore we do not attempt to perform such an analysis here. 5 However, we conclude this work by drawing attention to some interesting solutions that are of a different form than (46). These solutions are perhaps best illustrated by focusing on an algebra similar to the one described in (41). This algebra is defined by extending the KBc algebra with the two string fields In addition to the usual KBc commutation relations, the KLBB ′ c algebra satisfies Analytic solutions with the KLBB ′ c algebra can involve functions of the type F = F (K, L). It is important to note that this is a function of non-commuting variables. Therefore, some operations on F (K, L) will depend on how the function is ordered. In effort to state our results in the most convenient way, let us adopt the convention that we always order F (K, L) with every K appearing to the left of every L. In particular, the functions we will be interested in are those which can be written as First note that BL m = (L − 1) m B. Therefore, since B commutes with K, we have 6 It is similarly true that KF (K, L) = F (K, L − 1)K. Next we study the way B ′ interacts with F (K, L). Notice that since [[B ′ , K], K] = 0, we can use the formula Recalling the form of our function (49) and the rule (50), we find that B ′ satisfies the commutation relation The above equation raises an additional concern. Even with our prescribed ordering of the function F (K, L), there is still some confusion that may arise when taking the The above equation is actually quite intuitively pleasing. Since passing K through A(K, L) sends L → L − 1, it makes sense that passing ∂ ∂K through A(K, L) sends L → L + 1.
Recall the pure gauge ansatz U = 1 − F BcF . We obtain a new type of analytic solution by changing F (K) → F (K, L). Using the relationship (50), we find Notice, that the noncommutativity of K and L requires positioning the K and B factors appropriately on the two sides of the middle factor (1 − F 2 (K, L)) −1 . We postpone the detailed analysis of the physics of such solutions to a future work. Notice that we also have the freedom to consider a more general U of the form where F L i and F R i are both functions of the string fields K and L. The inverse of this pure gauge choice is given by The solution Ψ = UQU −1 looks somewhat more complicated because the summation prohibits some of our usual simplification tricks. However, it can still be written in the reasonably convenient form 7 This is a convenient form because the term Q(. . . ) will not contribute to a computation of the energy. By incorporating the new string field B ′ , we can consider a pure gauge ansatz U = 1 − F (K, L)B ′ cF (K, L). To efficiently compute U −1 , recall (52) and notice that 7 Similar solutions have been explored in [16].

Now we can compute
As usual, the corresponding solution is given by Ψ = UQU −1 . When dealing with solutions of the above type, one must be careful to use the rule (53) when computing the K derivative of a product of functions. One motivation for writing down these new solutions is in effort to construct solutions describing multiple D-brane configurations. Such an attempt has already been made in [5], but the solutions unfortunately failed some tests of regularity [6,7,8]. It is our hope that the extended KBc framework can be used to write down regular multibrane solutions. Also, it is apparent that some of these results can be extended to superstring field theory, following the work of [17,18].

Conclusion
We have constructed an interesting new representation of the zero central charge Virasoro algebra using string fields. We have used this construction to explore various extensions of the KBc algebra, and find new analytic solutions of open string field theory. It should be noted that many proposals have been made in the past which attempt to make use of left and right components. Some of these proposals are [19,20,21,22,23]. However, our work comes from a quite different perspective. We have been able to make insights not easily seen in previous constructions. The observations of this work are rich with opportunities for future exploration. Such exploration would include studying the surfaces generated by L n , computing the energy of the new solutions, and writing down a most general solution to the open string field theory equation of motion. This might necessitate revisiting and generalizing previous results, especially elucidating the role played by the so called hidden boundary [11,12].