D-brane Interactions in the IIA Plane-Wave Background

hep-th/040408 KAIST-TH 004/0 D-brane Interactions in the IIA Plane-Wave Background arxiv:hep-th/040408v 9 Jun 004 Yeonjung Kim, a and Jaemo Park b a Department of Physics, KAIST, Taejon 05-70, Korea b Department of Physics, POSTECH, Pohang 790-784, Korea Abstract We compute the D-brane tensions in the type IIA plane-wave background by comparing the interaction potential between widely separated D-branes in string theory with the supergravity mode exchange between the D-branes. We found that the D-brane tensions and RR charges in the plane-wave background are the same as those in the flat space. geni@muon.kaist.ac.kr jaemo@physics.postech.ac.kr

Introduction In a series of papers[],[],[],[4],[5],[6],[7], [8] simple type IIA string theory on the plane wave background have been studied, parallel to the development of the IIB string theory on the plane wave background [9],[0], [],[],[], [4]. The background for the string theory is obtained by compactifying the - dimensional plane wave background on a circle and taking the small radius limit. By working out the details of the resulting string theory one can obtain the useful information about the M-theory on the -dimensional plane wave background. However the resulting string theory in itself has many nice features and is worthy of the detailed study. It admits light cone gauge where the string theory spectrum is that of the free massive theory, which is similar to the IIB case. The world sheet enjoys (4,4) world sheet supersymmetry and the supersymmetry commutes with the Hamiltonian so that all members of the same supermultiplet has the same mass, which is different from the IIB theory. The various / BPS D-brane states were analyzed both in the light cone gauge and in the covariant formalism[],[]. Finally the boundary state formalism has developed in [],[7]. And the usual open-closed string channel duality was shown to hold for the supersymmetric D-brane configurations. As an application to this development, we work out the D-brane tensions and Ramond-Ramond (RR) charges in the IIA plane wave background. First we work out the open string partition function in the presence of widely separated D-branes. By taking a suitable limit, we find the contribution from the supergravity modes. By comparing this string theory computation with the corresponding supergravity calculation, we find that the supersymmetric D-brane tensions and RR charges are the same as those in the flat space. Similar result was obtained for the various IIB plane wave backgrounds []. In fact, we closely follow their approach in this paper. As explained in [], for the timelike branes, the result is more or less trivial. The interaction between a brane and an anti-brane is given by the overlap D p Dp where is the closed string propagator and Dp, D p are the corresponding boundary states. Due to the boundary condition, they satisfy p ˆ+ Dp = p ˆ+ D p = 0 where p ˆ+ is the light cone momentum operator. This condition projects the closed string propagator to the p ˆ+ = 0 subspace and these states propagate as in the flat space. However it is nontrivial to compute the tension of the space-like D-branes. Actual calculation shows that the supersymmetric D-brane tensions and RR charges are the same as those in flat space irrespective of their position in the flat space. In section, we present the string theory calculation for the interaction potential between two D-branes and in section we carry out the supergravity analysis. In the appendix, we provide the relevant information of the supergravity bulk action relevant for the calculation

in the text. String Theory Calculation The IIA plane wave background of our interest is given by ds = dx + dx A(x I )(dx + ) + 8 dx I dx I, (.) i= F + = µ, F +4 = µ (.) and A(x I ) = 4 i= µ 9 (Xi ) + 8 i =5 µ ) (.) 6 (Xi where X ± = (X 0 ± X 9 ). With the presence of the Ramond-Ramond background, the above plane wave background has SO() SO(4) where SO() acts on,, directions and SO(4) acts on 5,6,7,8 directions. We use the convention that unprimed coordinates denote,,,4 directions while primed coordinates denote 5,6,7,8 directions. For the worldsheet coordinates we use ± = ( τ ± σ ). The worldsheet action for the closed string theory is given by S LC = 4πα d σ( µ X + µ X + µ X I µ X I + m 9 4 i= X i X i + m 6 4 X i X i + b=±( iψ b +ψ b iψ b ψ b ) + im ψ + γ4 ψ im ψ γ4 ψ + ) (.4) i = where m = α p + µ and γ I are 8 8 matrices satisfying {γ I, γ J } = δ IJ. The sign of subscript ψ A ± denotes the eigenvalue of γ 4 while the superscript A =, denotes the eigenvalue of γ 9. The theory has two supermultiplets (X i, ψ, ψ + ),, ψ (Xi +, ψ ) of (4, 4) worldsheet supersymmetry with the mass m and m respectively. The fermions of the first supermultiplet 6 have γ 49 eigenvalue of while those of the second have the eigenvalue of. One can also consider the open strings with a suitable boundary conditions at the end of the open strings. One can use the same form of the action (.4) except for the interval for σ runs from 0 to π while for closed string σ runs from 0 to π. Possible supersymmetric boundary conditions or possible supersymmetric D-brane configurations were considered in [],[] and [7]. Corresponding boundary states were constructed in [] and [7]. For the spacelike branes, the possible type of supersymmetric D-brane configurations were tabulated in []. D0,D,D4,D6 spacelike branes are supersymmetric and one has to choose particular Neumann directions to satisfy the supersymmetric conditions. We first carry out the string theory calculation in the open string channel to get a correctly normalized amplitude and

extract the contribution from the lowest closed string modes. We then match these results with the supergravity calculation. As explained in [], in the standard light cone gauge X ± = α p + τ, X ± are automatically Neumann directions. Thus we will use the nonstandard light cone gauge for the open string X + = r+ π σ where r+ is the brane separation along the X + coordinate and σ is the worldsheet coordinate σ [0, π]. The Virasoro constraint determines X appearing in the string action is to be a Dirichlet direction as well. In this gauge, the mass parameter m = µr+ π. (.5) One subtle point when we work with the Lorentzian plane wave is that we are describing open strings in an inverted harmonic oscillator potential while the closed strings have the usual harmonic oscillator potential in the standard light cone[6]. It would be interesting to understand the full physical implication of the open strings in an inverted harmonic oscillator potential, which apparently could lead to negative norm states depending on the value of m, while in the closed string channel such potential pathologies do not appear. Some attempts to understand such subtleties were made in [6] The interaction energy between the branes can be written as E = i Tr( )Fs ln(l 0 iε) dt = i t Tr( )Fs e i(l 0 iε)t 0 (.6) where F s is the spacetime fermion number and the trace is taken over the open strings stretched between the branes and L 0 = p H lc with H lc being the light-cone Hamiltonian. We follow the convention of [] so that we work in the Lorentz signature for space time with a suitable ε prescription. For DpDp and DpD p branes separated in r +, r and the transversal x D, x D directions. dt f(x,x ) E = i 0 t e πit( 4π α ) ( sinh πtω 0 ) n N ( sinh πtω ) n N f iω 0 A (q)4 f iω 0 A (q)4 (.7) f iω 0 (q) 4 f iω 0 (q) 4 f(x, x ) = r + r + m r + sinm r +[(( x D ) + ( x D ) ) cosm r + x D x D ] m r + + sin m r +[(( x D ) + ( x D ) ) cosm r + x D x D ] (.8) where q = e πit and n N is the number of Neumann directions along 4 while n N is the number of those along 5678 with n N + n N = p +. Also m = µ, m = µ 6, ω 0 = m, ω 0 = m 6 while m is given by (.5).

The value A = for DpDp and A = 4 for DpD p configurations. while m, m are defined as f (m) (q) = q m ( q m ) / f (m) 4 (q) = q m m = (π) m = (π) ( q n= p= 0 ( q n +m ) n= (n ( ) p p= The modular transformation properties are given by ) +m ) (.9) ds e ps e π m s 0 ds e ps e π m s (.0) f m (e πit ) = f imt (e πi t ), f m 4 (e πit ) = f imt (e πi t ) (.) where f (m) (q) is defined by f (m) (q) = q m ( + q m ) / ( + q n +m ). The DpDp and DpD p brane configurations are aligned along the special directions which make the resulting Dp-brane configurations supersymmetric. One can see that in (.7), half of the contribution comes from one supermultiplet with the mass parameter m and the other half comes from the other supermultiplet with the mass parameter m. For the purpose of 6 calculating the tensions and RR charges of spacelike branes one can work out the region m, m < where open strings do not develop negative norm states. The large distance behavior of (.7) comes from the leading behavior of the integrand for small t. This is given by n= E Dp Dp E Dp D p = 4π(4π α ) p sin µr+ = 4π(4π α ) p cos µr+ sin µr+ 6 I9 p 0 (.) cos µr+ 6 I9 p 0 (.) where I 9 p 0 is the integrated propagator over (p + )-longitudinal directions with the separation in r +, r and the transverse directions for the associated propagator G 0 (x, x ) satisfying G 0 (x, x ) = iδ(x x ). This is given by 0 = i (iµr+ ) p (π) p 4 f(x, x ) p Γ( p) (µ ) n N ( µ 6 ) n N. (.4) sin µr+ sin µr+ 6 I 9 p 4

Field Theory Calculation We start from the type IIA supergravity action appeared in the appendix with D-brane source terms S p = T p d p+ x ge p 4 Φ + µ p A [p+] (.) where g stands for the induced metric on the worldvolume while T p and µ p are the brane tension and the RR charge of the D-brane in consideration. In the appendix, we obtain the gravity action to the quadratic order in the fluctuation around the plane wave background using the light-cone gauge. The resulting action is a sum of decoupled terms characterized by coefficients c and M S ψ = d 0 xψ α M ( iµc )ψ α. (.) In our case, ψ is in a tensor representation of SO() SO(4) and a contraction of tensor indices is understood. The details are explained in the appendix. The source terms contain the contribution of ψ α with ε = ± for brane/anti-brane respectively. S source = d 0 x δ 9 p (x x 0 ) k(ψ α + ǫ ψ α ). (.) The contribution of such a mode to the interaction is given by. D0-brane E = Mǫk cosµcr + I 9 p 0. (.4) We take the world volume direction to be X i = X. From the above source term (.), we have L source = it 0 (h φ) ± µ 0a. (.5) Using the notation of the appendix, this can be rewritten as L source = it 0 (h φ 0 8 (φ + φ ) 8 (φ 0 + φ 0 )) ± µ 0 4 (β + β + β 4 + β 4 ) (.6) where the definitions of the fields are given in the appendix. The value of M,k,c are summerized in the following table ψ h φ 0 φ (M, k, c) (4κ, it 0 4 ( κ, it 0 8 (64 9 κ, it 0 6 ψ φ 6 β β 4 (M, k, c) (64κ, it 0 6 µr+ ) (6κ, ±µ 0 4, µr+ (6κ, ±µ 0 4, µr+ ) 5

The sum of the contribution is given by [ E = κ I0 9 T0 + T 0 cosµr+ + ( T ] 0 µr+ µ 0 ) cos µr+ µ 0 cos comparing with the string result, we get (.7) T 0 = µ 0 = π κ (4π α ). (.8) Since we have SO() SO(4) symmetry, the same result would be obtained if D0-brane world voulume direction is X i with i=,,. This exhausts all the possible of the supersymmetry D- brane configurations. In the string theory analysis, we have the precisely the same condition for the supersymmetric D0-brane.. D brane According to the analysis in the string theory[5], the worldvolume directions of the supersymmetric D-brane can be taken to be (4) or (456) directions. The other configurations are equivalent to either of these by SO() SO(4) rotations. If we take the world volume direction to be (4), L source = it (h + h + h 44 φ) ± µ a 4 = it (h + h + φ 0 8 (φ + φ ) 8 (φ 0 + φ 0 )) ±µ 4 (β + β β 4 β 4 ) (.9) Again the contribution of the each field to the interaction energy is given by the table below. ψ h, h φ 0 φ (M, k, c) (4κ, it 4 ( κ, it 8 (64 9 κ, it 6 ψ φ 6 β β 4 (M, k, c) (64κ, it 6 µr+ ) (6κ, ±µ 4, µr+ (6κ, ±µ 4, µr+ ) The interaction energy is given by [ E = κ I0 7 T + T cosµr+ + ( T ] µr+ µ ) cos µr+ µ cos Again comparing with the string theory result, we get (.0) T = µ = 4π α (.) κ When the world volume direction of D-brane is 456, one can carry out similar computation, which gives the same values of T and µ. 6

. D4 brane If we take the world volume direction of the D4-brane to be (5678), then the coupling µ 4 A [5] = µ 4 d 5 x A 5678 = µ 4 d 5 x ε 4 5678A 4 (.) in the light cone gauge where ε i i i 8 is the totally antisymmetric tensor of rank 8. Thus the D4-brane in consideration is magnetically charged to the -form potential but for the computational purpose the contribution from (.) would be the same as in the D-brane case if we replace µ by µ 4. Thus we have to figure out the contribution from other remaining source terms. L source = it 4 (h + h 55 + h 66 + h 77 + h 88 + φ ) = it 4 (h + h 55 + h 66 + h 77 + h 88 φ 0 + 8 (φ 6 + φ 6 ) + 8 (φ + φ )) (.) The contribution of φ 0, φ, φ 6 are already worked out in D-brane case. Working out the contribution from the remaining gravitational sector we obtain the interaction energy [ E = κ I0 5 T4 + T 4 cosµr+ + ( T ] 4 µr+ µ 4 ) cos µr+ µ 4 cos. (.4) By the comparison with the string theory result, we get T 4 = µ 4 = π κ (4π α ). (.5) If the world volume direction is (78), we can work out the similar computation, which gives the same value of T 4 and µ 4. All the other supersymmetric D4-brane configurations are again related to the above two cases by SO() SO(4) rotations..4 D6 brane All supersymmetric configurations are equivalent to the D6-brane with world volume (45678). Again µ 6 [A 6 ] = µ 6 d 6 x a (.6) and we can borrow the computational result from the D0-brane. The other source terms are L source = it 6 ( i=45678 = it 6 ( i=5678 h ii + φ) h ii + φ 0 + 8 (φ + φ ) + 8 (φ 6 + φ 6 )). (.7) 7

By the similar calculation, one can obtain the interaction energy [ E = κ I0 T6 + T 6 cosµr+ + ( T ] 6 µ 6) cos µr+ µ 6 cos µr+. (.8) Thus T 6 = µ 6 = π κ (4π α ) (.9) to match the string theory computation. In conclusion, we find that for all supersymmetric Dp-branes of interest their tensions and charges are given by T p = µ p = π κ (4π α ) p. (.0) A Appendix In this appendix, we explain how to obtain the bulk action of the relavant field for the computation in the main text. In [5], the equations of motion for the IIA supergravity fluctuation to the leading order are obtained. They consists of the decoupled equation of motion of the form φ c + i µc φ c = 0 (A.) We use the leftmost subscript to indicate the coefficient c in the above equation in writing the various fields. The bosonic fields of IIA supergravity theory consist of the dilaton Φ, graviton g µν, one-form field A µ, two form field B µν and three form field potential A µνρ. We consider the small fluctuation of the above fields on the IIA plane wave background. Φ = φ g µν = ḡ µν + h µν A µ = Āµ + a µ B µν = b µν A µνρ = Āµνρ + a µνρ (A.) where ḡ µν, Ā µ and Āµνρ denote the IIA plane-wave background. We take the light cone gauge. a = b I = a IJ = h I = 0 (A.) Since the IIA plane-wave background has SO() SO(4) symmetry, it s convenient to classify the small fluctuations using this symmetry. SO() SO(4) scalar multiplets are given by φ 0 φ + h ii + h 44, φ φ + 4 ia 4 h 44, φ φ 4 ia 4 h 44, φ 6 φ 4ia h ii, φ6 φ + 4ia h ii. (A.4) 8

Here the subscript indicates the coefficient appearing in the mass parameter in the equaton of motion (A.). In the appendix, i denotes SO() direction while i denotes SO(4) one. For example, φ 6 satisfies φ 6 + iµ φ 6 = 0 (A.5) and its complex conjugate φ 6 satisfies φ 6 iµ φ6 = 0. (A.6) SO() vector multiplets are β 0i b 4i (A.7) β i a i ih 4i + i ǫ ijkb jk + ǫ ijk a 4jk, βi a i + ih 4i i ǫ ijkb jk + ǫ ijk a 4jk, β 4i a i + ih 4i + i ǫ ijkb jk ǫ ijk a 4jk, β4i a i ih 4i i ǫ ijkb jk ǫ ijk a 4jk Here again the leftmost subscript denotes the coefficient in the mass parameter. SO(4) vector multiplets are given by β i a i + ih 4i, βi a i ih 4i, β i b 4i i ǫ i j k l a j k l, βi b 4i + i ǫ i j k l a j k l (A.8) Then there are two index tensor fields. (ij) and (i j ) components are SO() and SO(4) graviton multiplets respectively. Thus we have h ij h ij δ ijh kk, h i j h i j 4 δ i j h k k (A.9) and the equations of motion are written as h ij = 0, h i j = 0 (A.0) And (ij ) components are defined by β ij b ij + i a 4ij, βij b ij i a 4ij, (A.) and (i j ) components are β i j a+ i j iã + i j, βi j a+ i j + iã + i j, β 4i j a i j + iã i j, β4i j a i j iã i j, (A.) where a ± i j b i j ± ǫ i j k l b k l, ã ± i j a 4i j ± ǫ i j k l a 4k l. 9

Finally we have two types of -rank tensor fields. (ijk ) components are β ijk a ijk iǫ ijkh kk, βijk a ijk + iǫ ijkh kk, (A.) while (ij k ) components are β 0ij k a ij k. (A.4) Consider the above diagonalized fields. One can obtain the action which gives the equation fo motion of each field. Since we started with the equation of motion, there are same ambiguities in the relative normalization of the fields. However such relative normalizations could be fixed by matching the gravity and the -form potential parts with the known form of the IIA actions in the light-cone gauge. The relavant part of the action needed for the computation in the main text is given by L = 8κ (h ij h ij + h i j h i j ) + κ φ 0 φ 0 + 9 64κ φ ( + iµ )φ + 64κ φ 6 ( + iµ )φ 6 + 6κ β i ( + iµ )β i + 6κ β 4i ( + 4iµ )β 4i + 8κ β i ( + iµ )β i + 6κ β i ( + iµ )β i + 6κ β ij ( + iµ )β ij + 64κ β iµ i j ( + )β i j + 64κ β 4iµ 4i j ( + )β 4i j + 6κ β ijk ( + iµ )β ijk + (A.5) where the omitted terms are not relevant for the computation in the main text. There are slight differences in the field definitions adopted here and in [5]. Our convention is that the coefficient in front of each field is consistent with the usual normalization of the p -form field p! 4κ d 0 x A [i i p] A [i i p] = 4κ The integrated propagator I 9 p c Acknowledgments d 0 x i <i < <i p A i i i p A i i i p. (A.6) (r +, r ) associated with (A.) is simply e icµr + I 9 p 0 (r +, r ). The work of J. P. and Y. K. is supported by the Korea Research Foundation (KRF) Grant KRF-00-070-C000. 0

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