Magnetically-enhanced open string pair production

We consider the stringy interaction between two parallel stacks of D3 branes placed at a separation. Each stack of D3 branes in a similar fashion carry an electric flux and a magnetic flux with the two sharing no common field strength index. The interaction amplitude has an imaginary part, giving rise to the Schwinger-like pair production of open strings. We find a significantly enhanced rate of this production when the two electric fluxes are almost identical and the brane separation is on the order of string scale. This enhancement will be largest if the two magnetic fluxes are opposite in direction. This novel enhancement results from the interplay of the non-perturbative Schwinger-type pair production due to the electric flux and the stringy tachyon due to the magnetic flux, and may have realistic physical applications.


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only to be non-vanishing but also to have an imaginary part. In general, the pair production rate is vanishing small and suppressed exponentially by the brane separation. So this pair production has no practical use even if string theories are relevant to our real world. However, when the magnetic fluxes are also present in a certain way, this open string pair production rate is greatly enhanced and becomes significant.
The purpose of this paper is to reveal this and to discuss its potential use and application. In section 2, we provide the basis for the computation of the real part of interaction amplitude for the system of two stacks of D3 branes with each stack carrying both electric and magnetic fluxes in a certain way. In section 3, we compute explicitly this amplitude and analyze the nature of the interaction. In section 4, we first analyze the small separation behavior of the amplitude computed in the previous section, then give the open string pair production rate and discuss its enhancement and significance. We conclude this paper in section 5.

The basic setup
In this section, we will provide the basis for computing the real part of the amplitude mentioned above. For this, we consider first the closed string cylinder digram with Dbranes represented by their respective boundary state |B [3][4][5][6]. For such a description, there are two sectors, namely NS-NS and R-R sectors. In each sector, we have two implementations for the boundary conditions of a D-brane, giving two boundary states |B, η , with η = ±. However, only the combinations |B NS = [|B, + NS − |B, − NS ] /2 and |B R = [|B, + R + |B, − R ] /2 are selected by the Gliozzi-Scherk-Olive (GSO) projection in NS-NS and R-R sectors, respectively. The boundary state |B, η for a Dpbrane can be expressed as the product of a matter part and a ghost part [7,8], i.e. |B, η = c p |B mat , η |B g , η /2 with |B mat , η = |B X |B ψ , η , |B g , η = |B gh |B sgh , η and the overall normalization As discussed in [9], the operator structure of the boundary state holds true even with the presence of external fluxes on the worldvolume and is always of the form |B X = exp(− ∞ n=1 1 n α −n · S ·α −n )|B X 0 and |B ψ , η NS = −i exp(iη ∞ m=1/2 ψ −m · S ·ψ −m )|0 for the NS-NS sector and |B ψ , η R = −exp(iη ∞ m=1 ψ −m · S ·ψ −m )|B, η 0R for the R-R sector. The ghost boundary states are the standard ones as given in [7], independent of the fluxes, which we will not present here. The matrix S and the zero-modes |B X 0 and |B, η 0R encode all information about the overlap equations that the string coordinates have to satisfy. They can be determined respectively [3][4][5]9] µ=0 |k µ = 0 for the bosonic sector, and |B ψ , η 0R = (CΓ 0 Γ 1 · · · Γ p 1+iηΓ 11 1+iη U ) AB |A |B for the R sector. In the above, the Greek indices α, β, · · · label the world-volume directions 0, 1, · · · , p along which the Dp brane extends, while the Latin indices i, j, · · · label the directions transverse to the brane, i.e., p + 1, · · · , 9. We defineF = 2πα F with F the external worldvolume field. We also have denoted by y i the positions of the D-brane along the transverse directions, by C the charge conjugation matrix and by U the matrix U (F ) = [− det(η+F )] −1/2 ; exp(−F αβ Γ α Γ β /2); with the symbol JHEP12(2017)076 ; ; denoting the indices of the Γ-matrices completely anti-symmetrized in each term of the exponential expansion. |A |B stands for the spinor vacuum of the R-R sector. Note that the η in the above denotes either sign ± or the worldvolume Minkowski flat metric and should be clear from the content.
The vacuum amplitude can be calculated via Γ = B(f 1 , g 1 )|D|B(f 2 , g 2 ) , where f a , g a with a = 1, 2 denote the corresponding electric and magnetic fluxes, and D is the closed string propagator defined as Here L 0 andL 0 are the respective left and right mover total zero-mode Virasoro generators of matter fields, ghosts and superghosts. For example, where L X 0 , L ψ 0 , L gh 0 and L sgh 0 represent contributions from matter fields X µ , matter fields ψ µ , ghosts b and c, and superghosts β and γ, respectively, and their explicit expressions can be found in any standard discussion of superstring theories, for example in [11], therefore will not be presented here. The above total vacuum amplitude has contributions from both NS-NS and R-R sectors, respectively, and can be written as Γ = Γ NSNS + Γ RR . In calculating either Γ NSNS or Γ RR , we need to keep in mind that the boundary state used should be the GSO projected one as given earlier. For this purpose, we need to calculate first the amplitude Γ(η , η) = B 1 , η |D|B 2 , η in each sector with η η = + or− and B a = B(f a , g a ).
In doing so, we can setL 0 = L 0 in the above propagator due to the fact thatL 0 |B = L 0 |B , which can be used to simplify the calculations. Given the structure of the boundary state, the amplitude Γ(η , η) can be factorized as where we have replaced the c p in the boundary state by nc p with n an integer to count the multiplicity of D p branes. In the above, we have In order to perform the calculations using the boundary states given earlier, we need to specify the D3 brane worldvolume gauge field.
The enhanced open string pair production rate occurs when we take, without loss of generality, the electric fluxF a 01 = −F a 10 = −f a with |f a | < 1, the magnetic fluxF a 23 = −F a 32 = −g a with |g a | < ∞, and the restF a αβ = 0. In other words, the electric flux and the magnetic one share no common field strength index. The corresponding matrix

The real part of the amplitude
Our computations of the real part of the amplitude follow [7,8,10]. With the preparation given in the previous section, the matrix elements in both NSNS and RR sectors can be JHEP12(2017)076 computed to give, for the ghosts, which are independent of the fluxes, while for matters, In the above, |z| = e −πt , V 4 denotes the D3 worldvolume, we have used the matrix S property (S T ) µ ρ S ρ ν = δ µ ν to simplify the computations, and .

JHEP12(2017)076
Here we have defined λ = e 2πiν , λ = e 2πiν and used This amplitude can be expressed nicely in terms of θ-functions and the Dedekind η-function with their standard definitions as given, for example, in [13] and is where the following identity has been used which is a special case of more general identity given in [14]. In (3.8), we have set ν = iν 0 with 0 < ν 0 < ∞ and ν = ν 0 with 0 < ν 0 < 1 and in terms of ν 0 and ν 0 , we have , , cos πν 0 = 1 + g 1 g 2 (1 + g 2 1 )(1 + g 2 2 ) , , where |f a | < 1 and |g a | < ∞ (a = 1, 2). The amplitude (3.8) can be further expressed as where we have used the explicit expressions for θ 1 (ν|τ ) and η(τ ) and The large y amplitude comes from the large t integration for which D n ≈ 1 and can be checked to give the expected attractive interaction (Γ > 0). The small t contribution to the amplitude becomes important only for small y. The numerator and the factor in the denominator, (1 − 2|z| 2n cos πν 0 + |z| 4n ) > (1 − |z| 2n ) 2 , in D n are both positive while the factor (1 − 2|z| 2n cosh 2πν 0 + |z| 4n ) in the denominator is positive for large t but it can be negative for small enough t. Therefore the nature of the small y interaction (attractive or repulsive) is unclear in terms of the integration variable t since the infinite product involves an infinite number of such factors even if each of them is negative in the integrand. So we expect some interesting physics to appear for small y.

JHEP12(2017)076 4 The enhanced open string pair production
The appropriate frame for exploring the small y physics and the analytic structure of the amplitude (3.11) in the short cylinder limit t → 0 is in terms of the annulus variable t of opens string description. This can be achieved via the Jacobi transformation t → t = 1/t. So in terms of the annulus variable t , noting η(τ ) = η(−1/τ )/(−iτ ) 1/2 and θ 1 (ν|τ ) = ie −iπν 2 /τ θ 1 (ν/τ | − 1/τ )/(−iτ ) 1/2 , we can re-express the amplitude (3.11) as where in the second equality we have dropped the prime on t and .

(4.2)
In the above, |z| = e −πt and for n ≥ 1, E n > 0 since 0 < ν 0 < 1. The amplitude vanishes when f 1 = f 2 and g 1 = g 2 and this has to be true since the underlying system is just like each stack of the D3 branes, preserving one half of spacetime supersymmetry. The factor sin πν 0 t in the integrand of (4.1) once again makes it unclear about the nature of the interaction though all other ones are positive for 0 < t < ∞. In spite of this, we do have a new feature showing up. Note that this factor sin πν 0 t vanishes at t k = k/ν 0 with k = 1, 2, · · · and the integrand blows up at these points. So we have an infinite number of simple poles of the integrand and the natural interpretation of these simple poles are the creations of various open string pairs due to the electric flux [15,16], the analog of Schwinger pair production in QED. The rate of open string pair production per unit worldvolume is the imaginary part of the amplitude, which can be obtained as the sum of the residues of the poles of the integrand in (4.1) times π following [15,16] and is given as (4.4) We come now to examine various instabilities. First for large t in (4.1) or large k in (4.3), there is a divergent factor exp[−t(y 2 − 2π 2 ν 0 α )/(2πα )] or exp[−k(y 2 − 2π 2 ν 0 α )/(2πν 0 α )] when y < π 2ν 0 α , signaling the onset of tachyonic instability [17,18]. This instability is due to the presence of magnetic fluxes. So the computations of the amplitude Γ and JHEP12(2017)076 the rate W are valid only for y ≥ π 2ν 0 α [19,20]. For the two electric fluxes, we can set f a = 1 − a with a ≥ 0. Their respective critical value corresponds to set a → 0. When either or both approach their respective critical values but keeping 1 / 2 → 0 or ∞, we have ν 0 → ∞ from the first two equations in (3.10) and expect the pair production rate (4.3) to diverge. One can easily check that this is indeed true using (4.3) and (4.4). The above instabilities are expected. For small enough ν 0 and a fixed non-vanishing ν 0 such that ν 0 /ν 0 1, the rate (4.3) becomes where we have used F k,n ≈ 1. It is clear from (4.5) that when |g 1 | and |g 2 | are fixed, the largest rate (also largest ν 0 ) occurs when the two fluxes are opposite in direction. From (3.10), small enough ν 0 implies small enough |f 1 − f 2 |. This further implies that the two electric fluxes are almost identical. A very special case of g 1 = f 2 = 0 was considered before by the present author and his collaborator in [21]. This corresponds to a system of one stack of branes carrying an electric flux and the other stack carrying a magnetic flux. The small enough ν 0 gives there |f 1 | 1 which is much less generic than the present |f 1 − f 2 | 1 since in the same physical environment the magnitude of electric flux carried by any stack of branes should not be much different and is less than unity but cannot be too small in general. The condition |f 1 | 1 considered in [21] is for academic purpose but quite unnatural in practice. In other words, the present condition |f 1 − f 2 | 1 is more useful and more suitable for potentially realistic applications discussed later in section 5.
We now compare the rate (4.5) to the one with the same ν 0 but without the magnetic fluxes as given in [10]. This latter rate can also be obtained from (4.3) via the limits of g a = 0, ν 0 = 0 as where we have set k = 2l − 1 and the even k doesn't contribute to this rate. So it is clear for each odd k = 2l − 1, there is a greatly enhanced factor where the superscript 'l' denotes the l-th term in the corresponding rate summation. For small enough ν 0 and reasonable large magnetic flux, this enhancement can be very significant. Now the corresponding rate can be approximated by the first term k = 1 or l = 1 and the enhancement factor is |g 1 − g 2 |e πν 0 /ν 0 /4ν 0 . Let us make a sample numerical estimation of this enhancement to demonstrate its significance. It has a value of 3.2 × 10 35 , a very significant enhancement, for ν 0 = 0.02, ν 0 = 0.5. This can be achieved using (3.10) via a moderate choice of g 1 = −g 2 = 1 (noting |g a | < ∞) and f 1 = 0.2 with f 2 = f 1 − and |f 1 − f 2 | = | | ≈ πν 0 (1 − f 2 1 ) = 0.06 1. To be physically significant, we need the rate JHEP12(2017)076 itself in string units to be large enough, not merely the enhancement factor. The rate in string units for the above sample case can be estimated to be with a typical choice of n 1 = n 2 = 10. So this rate (2πα ) 2 W(ν 0 = 0.5) = 0.61, quite significant, at y = π √ α + 0 + ≈ π √ α , a few times of string scale and before the onset of tachyon condensation, but decreases exponentially with the separation y 2 for y > π √ α . For example, the rate becomes half of its maximal value at y − π √ α ≈ 0.01 √ α , just 1% of the string scale. The similar rate for a general p ≥ 3 in string units can be computed to give 2 which gives the rate for p > 3 smaller than that for p = 3 by at least a factor of (ν 0 /4π) 1/2 ≈ 0.04 for the above sample case. So for the case of branes carrying one electric flux and one magnetic flux, the largest rate is for p = 3 and the rate for the other branes with p > 3 is at least one order of magnitude smaller given the fact that ν 0 /ν 0 1 and ν 0 < 1.

Conclusion and discussion
It is clear by now that the open string pair production enhancement comes from the interplay of the non-perturbative Schwinger-type pair production due to the presence of the electric flux and the stringy tachyon due to that of the magnetic flux. This enhanced rate can be significant for a brane separation of a few times of string scale and before the onset of tachyon condensation. This may have potentially realistic observational consequences. An electric flux can give rise to the Schwinger-type pair production and an additional magnetic flux can enhance this effect even for an isolated stack of branes carrying these fluxes [22,23]. In general, this pair production is too small to be detected. However, the enhanced pair production discussed in this paper is quite different and purely stringy, and results from two stacks of branes with each carrying the electric and magnetic fluxes. This production is very sensitive to the brane separation as described above. An observer on one stack of branes, though unable to sense the other stack directly, may detect a significant increase of pair production when the other stack of branes come at separation of the order of string scale. This is purely stringy and therefore provides a means to detect the existence of extra dimensions and also a test of this theory. This type of enhanced pair production occurs only for p ≥ 3 and the largest rate is for p = 3 (at least one order smaller for p > 3). So this detection can single out D3 branes as the most preferable to its observer, if he/she just like us knows about string theory. The produced large number of open string pairs can in turn annihilate to give, for example, highly concentrated high energy photons if the fluxes are localized on the branes and this may have observational consequence such as the Gamma-ray burst. This pair production and its subsequent annihilation may also useful in providing a new mechanism for reheating process after cosmic inflation.