1008/1008.2430.md

Conductivity at finite 't Hooft coupling from AdS/CFT

M. Ali-Akbari¹ and K. Bitaghsir Fadafan²

¹School of Physics, Institute for Research in Fundamental Sciences (IPM)
P.O.Box 19395-5531, Tehran, Iran

E-mails: aliakbari@theory.ipm.ac.ir

²Physics Department, Shahrood University of Technology,
P.O.Box 3619995161, Shahrood, Iran

E-mails: bitaghsir@shahroodut.ac.ir

Abstract

We use the AdS/CFT correspondence to study the DC conductivity of massive $\mathcal{N} = 2$ hypermultiplet fields in an $\mathcal{N} = 4$ $SU(N_c)$ super-Yang-Mills theory plasma in the large $N_c$ and finite 't Hooft coupling. We also discuss general curvature-squared and Gauss-Bonnet corrections on the DC conductivity.# Contents

1	Introduction	2
2	Review of conductivity	4
3	$\backslash mathcal\{R\}^4$ corrections to AdS-Schwarzschild black brane	6
3.1	Ohmic conductivity . . . . .	7
3.2	Conductivities in the presence of magnetic field . . . . .	8
4	$\backslash mathcal\{R\}^2$ corrections to AdS-Schwarzschild black brane	10
5	Discussion and Conclusion	15

1 Introduction

Anti-de Sitter/conformal field theory correspondence (AdS/CFT) conjectures that IIB string theory on $AdS_5 \times S^5$ background is dual to $D = 4$ $\mathcal{N} = 4$ $SU(N_c)$ super Yang-Mills theory (SYM) [1]. In the limits of large $N_c$ and large 't Hooft coupling $\lambda = g_{YM}N_c^2$ , the SYM theory is dual to IIB supergravity which is low energy effective theory of superstring theory. As a result a thermal SYM theory corresponds to supergravity in an AdS-Schwarzschild background where the SYM theory temperature is identified with the Hawking temperature of the AdS black hole [2].

AdS/CFT idea has been applied to study different aspects of strongly coupled SYM theory. Recently the application of this duality in condensed matter physics (called AdS/CMT) has been studied [3]. This duality is very useful to study certain strongly coupled systems in CMT by holography techniques and to understand better their properties. A quantity attracting attentions and computing is conductivity [4]. In order to compute conductivity, it is necessary to add spinor fields in fundamental representation. As it is well-known fields in the $\mathcal{N} = 4$ SYM theory are in adjoint representation and by introducing $\mathcal{N} = 2$ hypermultiplets one can include fields in the fundamental representation. To do so on gravity side, $N_f$ flavor branes are introduced in the probe limit meaning we have only $N_f \ll N_c$ of them and the AdS background is left unchanged. In other words, open string degrees of freedom are now considered. On the gauge theory side this corresponds to $\mathcal{N} = 2$ supersymmetric hypermultiplet flavor fields propagatingin SYM theory. The local $U(N_f)$ symmetry on the D7-branes corresponds to global $U(N_f)$ symmetry whose $U(1)_B$ subgroup may be identified with baryon number. Non-dynamical electric and magnetic fields can be coupled to $U(1)B$ charge and we then expect a constant, nonzero currents. Hence the conductivity tensor $\sigma{ij}$ is identified by

$$⟨J_i⟩={\sigma }_{ij}{E}_j\mathrm{.}(1)\backslash langle\; J\_i\; \backslash rangle\; =\; \backslash sigma\_\{ij\}\; E\_j.\; \backslash quad\; (1)$$

Electric and magnetic fields produce diagonal and off-diagonal elements in conductivity tensor respectively. In fact on the gravity side currents, electric and magnetic fields are introduced as nontrivial gauge fields living on the D7-branes.

The DC conductivity in "strange metals" has been studied in [7, 8]. It was found that conductivity is independent of the dimensionality of a probe brane in the background created by a stack of $D_p$ -branes [6]. Also it was shown that the properties of the DC conductivity can be studied by that of the single heavy quark. One should consider massive carriers as endpoint of strings which end on flavor branes and use the quasi-particle description. Then it would be straightforward to calculate the DC conductivity from the drag force calculations[8, 9]. We discuss this approach in the last section.

In this paper we study higher derivative corrections on the DC conductivity. These corrections on the gravity side correspond to finite coupling corrections on the gauge theory side. The main motivation to consider corrections comes from the fact that string theory contains higher derivative corrections arising from stringy effects. In the case of $\mathcal{N} = 4$ SYM theory, the leading order correction in $1/\lambda$ arises from stringy correction to the low energy effective action of type IIb supergravity, $\alpha'^3 \mathcal{R}^4$ . We study $\mathcal{R}^4$ and $\mathcal{R}^2$ corrections to the DC conductivity. An understanding of how these computations are affected by finite $\lambda$ corrections may be essential for more precise theoretical predictions.

The article is organized as follows. In the next section, we will give a brief review of [4, 5] and then follow the same direction and study Ohmic and Hall conductivities in the presence of corrections in section 3. Moreover in section 4, we consider general $\mathcal{R}^2$ and Gauss-Bonnet corrections and in the last section we draw our conclusions and summarize our results.## 2 Review of conductivity

In this section we will give a brief review of [4, 5]. The AdS-Schwarchild metric, in units where the radius of $AdS$ is one, is ¹

$$d{s}^2=G_{tt}d{t}^2+G_{xx}d{\vec{x}}^2+G_{uu}d{u}^2+d^2{\mathrm{\Omega }}_5\mathrm{.}(2)ds^2\; =\; G\_\{tt\}\; dt^2\; +\; G\_\{xx\}\; d\backslash vec\{x\}^2\; +\; G\_\{uu\}\; du^2\; +\; d^2\backslash Omega\_5.\; \backslash quad\; (2)$$

Here $d\vec{x}^2$ is the three dimensional space and the metric functions are given by

$$G_{tt}=-u^2(1-\frac{u_0^4}{u^4}),(3a)G\_\{tt\}\; =\; -u^2(1\; -\; \backslash frac\{u\_0^4\}\{u^4\}),\; \backslash quad\; (3a)$$

$$G_{xx}=u^2,(3b)G\_\{xx\}\; =\; u^2,\; \backslash quad\; (3b)$$

$$G_{uu}=u^{-2}(1-\frac{u_0^4}{u^4}{)}^{-1},(3c)G\_\{uu\}\; =\; u^\{-2\}(1\; -\; \backslash frac\{u\_0^4\}\{u^4\})^\{-1\},\; \backslash quad\; (3c)$$

where $u_0$ is event horizon. Also $S^5$ metric is

$$d{\mathrm{\Omega }}_5^2=d{\theta }^2+{\sin }^2\theta d{\psi }^2+{\cos }^2{\theta }^{2}d{\mathrm{\Omega }}_3^2\mathrm{.}(4)d\backslash Omega\_5^2\; =\; d\backslash theta^2\; +\; \backslash sin^2\backslash theta\; d\backslash psi^2\; +\; \backslash cos^2\backslash theta^2\; d\backslash Omega\_3^2.\; \backslash quad\; (4)$$

where $d\Omega_3^2$ is the metric of $S^3$ and $\theta$ runs from zero to $\frac{\pi}{2}$ . In addition the Hawking temperature is given by

$$T=\frac{u_0}{\pi }\mathrm{.}(5)T\; =\; \backslash frac\{u\_0\}\{\backslash pi\}.\; \backslash quad\; (5)$$

In order to find conductivity a number $N_f$ of D7-branes filling $AdS_5$ and wrapping the $S^3 \subset S^5$ have been considered in the AdS-Schwarchild background. Moreover worldvolume gauge fields $A_t(u)$ , $A_x(u, t) = -Et + f_x(u)$ and $A_y(u, t) = Bx + f_y(u)$ as well as the $\theta(u)$ describing the position $S^3$ on the $S^5$ are turned on. The above system is described by Dirac-Born-Infeld action. From the gauge field equations of motion, conserved charges $Q$ , $I^x$ and $I^y$ associated with $A_t(u)$ , $A_x(u, t)$ and $A_y(u, t)$ are found. The conserved charges which are sub-leading, normalizable terms of asymptotic expansion can be related to expectation value of dual operators i.e.

$$⟨J^t⟩=Q,⟨J^x⟩=I^x,⟨J^y⟩=I^y\mathrm{.}(6)\backslash langle\; J^t\; \backslash rangle\; =\; Q,\; \backslash quad\; \backslash langle\; J^x\; \backslash rangle\; =\; I^x,\; \backslash quad\; \backslash langle\; J^y\; \backslash rangle\; =\; I^y.\; \backslash quad\; (6)$$

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¹A change of variable as $uz = 1 + \frac{z^4}{u^4}$ relates our coordinate to what is used in [4].Having worked out the gauge fields in terms of $Q$ and $B$ one can write the on-shell action as follows [5]

$$S_{D7}=-{\mathcal{N}}^2(2\pi {\alpha }^{\mathrm{\prime }}{)}^2\int d^{4}x{\cos }^6\theta g_{xx}^2\sqrt{g_{tt}{g}_{uu}}\frac{\xi }{\sqrt{\xi \chi -a^2}},(7)S\_\{D7\}\; =\; -\backslash mathcal\{N\}^2(2\backslash pi\backslash alpha\text{'})^2\; \backslash int\; d^4x\; \backslash cos^6\backslash theta\; g\_\{xx\}^2\; \backslash sqrt\{g\_\{tt\}g\_\{uu\}\}\; \backslash frac\{\backslash xi\}\{\backslash sqrt\{\backslash xi\backslash chi\; -\; a^2\}\},\; \backslash quad\; (7)$$

where $\mathcal{N} = \frac{\lambda}{(2\pi^4)} N_f N_c$ . $g_{tt}(= |g_{tt}|)$ , $g_{uu}$ and $g_{xx}$ are components of induced metric and

$$\xi =g_{tt}{g}_{xx}^2+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2(g_{tt}{B}^2-g_{xx}{E}^2),(8a)\backslash xi\; =\; g\_\{tt\}g\_\{xx\}^2\; +\; (2\backslash pi\backslash alpha\text{'})^2(g\_\{tt\}B^2\; -\; g\_\{xx\}E^2),\; \backslash quad\; (8a)$$

$$\chi =g_{tt}{g}_{xx}^2({\mathcal{N}}^2(2\pi {\alpha }^{\mathrm{\prime }}{)}^4{g}_{xx}{\cos }^6\theta )+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2(g_{tt}{Q}^2-g_{xx}(I_x^2+I_y^2)),(8b)\backslash chi\; =\; g\_\{tt\}g\_\{xx\}^2\; (\backslash mathcal\{N\}^2(2\backslash pi\backslash alpha\text{'})^4\; g\_\{xx\}\; \backslash cos^6\backslash theta)\; +\; (2\backslash pi\backslash alpha\text{'})^2\; (g\_\{tt\}Q^2\; -\; g\_\{xx\}(I\_x^2\; +\; I\_y^2)),\; \backslash quad\; (8b)$$

$$a=(2\pi {\alpha }^{\mathrm{\prime }}{)}^2(g_{tt}{I}^{x}B+g_{xx}{I}^{y}E)\mathrm{.}(8c)a\; =\; (2\backslash pi\backslash alpha\text{'})^2\; (g\_\{tt\}I^x\; B\; +\; g\_\{xx\}I^y\; E).\; \backslash quad\; (8c)$$

$\xi$ , as a function of $u$ , has negative and positive value at the horizon and near the boundary respectively. In fact at a specific point, say $u_*$ , we have $\xi(u_*) = 0$ . Hence $u_*$ is

$$u_{\ast }^4=u_0^4\mathcal{F}(e,b)={\pi }^4{T}^4\mathcal{F}(e,b)=g_{xx}^2(u_{\ast })(9)u\_*^4\; =\; u\_0^4\; \backslash mathcal\{F\}(e,\; b)\; =\; \backslash pi^4\; T^4\; \backslash mathcal\{F\}(e,\; b)\; =\; g\_\{xx\}^2(u\_*)\; \backslash quad\; (9)$$

where²

Reality condition of $\sqrt{\xi\chi - a^2}$ imposes that two functions $\chi$ and $a$ must vanish at $u = u_*$ . By setting (8b) and (8c) to zero at $u_*$ and converting to field theory quantities, Ohmic and Hall conductivities become

$${\sigma }_{xx}=\sqrt{\frac{N_f^2{N}_c^2{\cos }^6{\theta }_{\ast }{\mathcal{F}}^{3\mathrm{/}2}}{16{\pi }^2(b^2+\mathcal{F})}{T}^2+\frac{q^2\mathcal{F}}{(b^2+\mathcal{F}{)}^2}}(11a)\backslash sigma\_\{xx\}\; =\; \backslash sqrt\{\backslash frac\{N\_f^2\; N\_c^2\; \backslash cos^6\; \backslash theta\_*\; \backslash mathcal\{F\}^\{3/2\}\}\{16\backslash pi^2\; (b^2\; +\; \backslash mathcal\{F\})\}\; T^2\; +\; \backslash frac\{q^2\; \backslash mathcal\{F\}\}\{(b^2\; +\; \backslash mathcal\{F\})^2\}\}\; \backslash quad\; (11a)$$

$${\sigma }_{xy}=\frac{qb}{b^2+\mathcal{F}}(11b)\backslash sigma\_\{xy\}\; =\; \backslash frac\{qb\}\{b^2\; +\; \backslash mathcal\{F\}\}\; \backslash quad\; (11b)$$

The Ohmic conductivity depends on magnetic field, electric field and the temperature of the field theory, simplicity we name it as $\sigma(B, E, T)$ . This quantity has two main terms

$${\sigma }_{xx}(B,E,T)=\sqrt{{\widehat{\sigma }}_0^2+{\widehat{\sigma }}^2}(12)\backslash sigma\_\{xx\}(B,\; E,\; T)\; =\; \backslash sqrt\{\backslash hat\{\backslash sigma\}\_0^2\; +\; \backslash hat\{\backslash sigma\}^2\}\; \backslash quad\; (12)$$

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²Notice that $\alpha'^{-2} = 4\pi g_s N_c = g_{YM}^2 N_c = \lambda$ .where $\hat{\sigma}_0$ arises from thermally produced pairs of charge carriers. By increasing the mass of carriers, $\hat{\sigma}_0$ can be made arbitrary small and the leading term in conductivity will be $\hat{\sigma}$ . This term can be found by studying the properties of a moving single string and calculating drag force [4]. We will discuss this point in the discussion section.

In next section we will follow the same direction and study above conductivities in the presence of correction.

3 $\mathcal{R}^4$ corrections to AdS-Schwarzschild black brane

Since $AdS/CFT$ correspondence refers to complete string theory, one should consider the string corrections to the 10D supergravity action. The first correction occurs at order $(\alpha')^3$ [13]. In the extremal $AdS_5 \times S^5$ it is clear that the metric does not change [14], conversely this is no longer true in the non-extremal case. Corrections in inverse 't Hooft coupling $1/\lambda$ which correspond to $\alpha'$ corrections on the string theory side were found in [13]. Higher derivative corrections i.e. $\mathcal{R}^2$ and $\mathcal{R}^4$ on the rotating quark-antiquark system in the hot plasma and on the drag force on a moving heavy quark have been investigated in [10, 11, 12].

Functions of the $\alpha'$ -corrected metric are given by [15]

where

and $w = \frac{u}{u_0}$ . There is an event horizon at $u = u_0$ and the geometry is asymptotically $AdS$ at large $u$ with a radius of curvature $R = 1$ . The expansionparameter $k$ can be expressed in terms of the inverse 't Hooft coupling as

$$k=\frac{\zeta (3)}{8}{\lambda }^{-3\mathrm{/}2}\sim 0.15{\lambda }^{-3\mathrm{/}2}\mathrm{.}(15)k\; =\; \backslash frac\{\backslash zeta(3)\}\{8\}\; \backslash lambda^\{-3/2\}\; \backslash sim\; 0.15\; \backslash lambda^\{-3/2\}.\; \backslash quad\; (15)$$

The temperature is given by

$$T_{{\mathcal{R}}^4}=\frac{u_0}{\pi (1-k)}\mathrm{.}(16)T\_\{\backslash mathcal\{R\}^4\}\; =\; \backslash frac\{u\_0\}\{\backslash pi(1-k)\}.\; \backslash quad\; (16)$$

In order to find conductivities we set all of equations (8) to zero where the induced metric components will now be computed by (13).

3.1 Ohmic conductivity

Here we focus on a case where the magnetic field has been turned off and (8a), after setting to zero, becomes

$$w^{16}-(1+75k+e^2)w^{12}-k(\frac{25}{8}{w}^8-120w^4+\frac{335}{8})=0,(17)w^\{16\}\; -\; (1\; +\; 75k\; +\; e^2)w^\{12\}\; -\; k\; \backslash left(\; \backslash frac\{25\}\{8\}w^8\; -\; 120w^4\; +\; \backslash frac\{335\}\{8\}\; \backslash right)\; =\; 0,\; \backslash quad\; (17)$$

up to first order in $k$ perturbatively. $u_* = u_0 w_*$ is a real parameter and takes value between $u_0$ and infinity. These two conditions tell us that just a root of (17) is acceptable for $w_*$ among sixteen roots. Now (8b) and (8c) must be set to zero. (8c) leads to $I^y = 0$ and (8b) becomes

$${\sigma }_{xx}=\frac{I^x}{E}=\sqrt{{\mathcal{N}}^2(2\pi {\alpha }^{\mathrm{\prime }}{)}^4{g}_{xx}{\cos }^6{\theta }_{\ast }+\frac{(2\pi {\alpha }^{\mathrm{\prime }}{)}^2}{g_{xx}^2}{Q}^2}\mathrm{.}(18)\backslash sigma\_\{xx\}\; =\; \backslash frac\{I^x\}\{E\}\; =\; \backslash sqrt\{\backslash mathcal\{N\}^2\; (2\backslash pi\backslash alpha\text{'})^4\; g\_\{xx\}\; \backslash cos^6\; \backslash theta\_*\; +\; \backslash frac\{(2\backslash pi\backslash alpha\text{'})^2\}\{g\_\{xx\}^2\}\; Q^2\}.\; \backslash quad\; (18)$$

where $g_{xx}$ evaluated at $u_*$ , which is found by solving (17), is given by

$$g_{xx}(u_{\ast })={\pi }^2{T}^2(\sqrt{1+e^2}+\frac{5k(-10+e^2(163+120e^2(3+e^2)))}{16(1+e^2{)}^{7\mathrm{/}2}}),(19)g\_\{xx\}(u\_*)\; =\; \backslash pi^2\; T^2\; \backslash left(\; \backslash sqrt\{1\; +\; e^2\}\; +\; \backslash frac\{5k(-10\; +\; e^2(163\; +\; 120e^2(3\; +\; e^2)))\}\{16(1\; +\; e^2)^\{7/2\}\}\; \backslash right),\; \backslash quad\; (19)$$

Finally by substituting (19) in (18) the Ohmic conductivity becomes

where

$${\sigma }_{xx}^{\mathcal{N}=4}=\sqrt{\frac{N_f^2{N}_c^2{T}^2}{16{\pi }^2}\sqrt{1+e^2}{\cos }^6{\theta }_{\ast }+\frac{q^2}{1+e^2}}\mathrm{.}(21)\backslash sigma\_\{xx\}^\{\backslash mathcal\{N\}=4\}\; =\; \backslash sqrt\{\backslash frac\{N\_f^2\; N\_c^2\; T^2\}\{16\backslash pi^2\}\; \backslash sqrt\{1\; +\; e^2\}\; \backslash cos^6\; \backslash theta\_*\; +\; \backslash frac\{q^2\}\{1\; +\; e^2\}\}.\; \backslash quad\; (21)$$

We would like to emphasize two points about our result. First, at finite temperature for a large value of electric field second term in the conductivity equation coming from correction goes to zero which means that correction of metric is negligible. Second, depending on other parameters, conductivity increases, decreases or does not change. In particular by taking large mass limit $\cos \theta_* \rightarrow 0$ [1, 2] there is a critical value of electric field $e_c = 0.233745$ where the correction effect vanishes. As a result conductivity increases when $e < e_c$ and vice versa. In the limit of zero density, if $e > e_c$ or $e < e_c$ we have a positive or negative correction effect, respectively.

3.2 Conductivities in the presence of magnetic field

In this section, we study the effect of 't Hooft coupling correction on the conductivities when the magnetic field is turned on. In order to do that by setting (8) to zero, we have

$$w(w-1)(16w^3-1200k{w}^2-1275kw+645k)+e^{2}w(-16w^3+25kw+25k)(22a)w(w\; -\; 1)(16w^3\; -\; 1200kw^2\; -\; 1275kw\; +\; 645k)\; +\; e^2w(-16w^3\; +\; 25kw\; +\; 25k)\; \backslash quad\; (22a)$$

$$+b^2(w-1)(16w^3-1200k{w}^2-1225kw+695k)=0,{\sigma }_{xx}=\frac{g_{xx}}{g_{xx}^2+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2{B}^2}\sqrt{(2\pi {\alpha }^{\mathrm{\prime }}{)}^4\mathcal{N}(g_{xx}^2+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2{B}^2)g_{xx}{\cos }^6{\theta }_{\ast }+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2{Q}^2},(22b)+\; b^2(w\; -\; 1)(16w^3\; -\; 1200kw^2\; -\; 1225kw\; +\; 695k)\; =\; 0,\; \backslash \backslash \; \backslash sigma\_\{xx\}\; =\; \backslash frac\{g\_\{xx\}\}\{g\_\{xx\}^2\; +\; (2\backslash pi\backslash alpha\text{'})^2\; B^2\}\; \backslash sqrt\{(2\backslash pi\backslash alpha\text{'})^4\; \backslash mathcal\{N\}(g\_\{xx\}^2\; +\; (2\backslash pi\backslash alpha\text{'})^2\; B^2)\; g\_\{xx\}\; \backslash cos^6\; \backslash theta\_*\; +\; (2\backslash pi\backslash alpha\text{'})^2\; Q^2\},\; \backslash quad\; (22b)$$

$${\sigma }_{xy}=\frac{(2\pi {\alpha }^{\mathrm{\prime }}{)}^{2}QB}{g_{xx}^2+(2\pi {\alpha }^{\mathrm{\prime }}{)}^2{B}^2}\mathrm{.}(22c)\backslash sigma\_\{xy\}\; =\; \backslash frac\{(2\backslash pi\backslash alpha\text{'})^2\; QB\}\{g\_\{xx\}^2\; +\; (2\backslash pi\backslash alpha\text{'})^2\; B^2\}.\; \backslash quad\; (22c)$$

where as before $g_{xx}$ and $\cos \theta$ in (22b) and (22c) are evaluated at $w = w_*$ . In this case $w_*$ will be found by solving (22a). However this equation is complicated one can solve it numerically. We assume different values for parameters and discuss behavior of Ohmic and Hall conductivities in terms of them. In the massive case, $\cos \theta \rightarrow 0$ , we have plotted conductivities versus $e$ and $b$ in Fig. 1-4. Our figures have been plotted at fixed temperature( $u_0 = 3$ ) and for three different values of $k(=0.0001, 0.001, 0.01)$ .Ohmic conductivity has been plotted in Fig. 1. In the left plot of this figure $b = 10$ . Notice that from (15), increasing $k$ corresponds to decreasing 't Hooft coupling constant $\lambda$ . For small values of $\lambda$ , there is a specific maximum value for Ohmic conductivity. It is clearly seen that by increasing 't Hooft coupling constant the shape of Ohmic conductivity changes and it approximately starts from its maximum value. In the right plot of Fig. 1 $b = 30$ . As one finds from (22), by increasing $b$ the value of Ohmic conductivity will be decreased. This behavior of Ohmic conductivity is clearly shown in this plot. In addition by increasing $b$ , the maximum value of Ohmic conductivity appears at larger value of $e$ .

Figure 1: $\sigma_{xx}$ versus $e$ for different values of $k$ at fixed $b$ . Left: $b = 10$ . Right: $b = 30$ .

It would also be interesting to investigate behavior of Ohmic conductivity in terms of $b$ at constant $e$ . In the left and right plots of Fig 2, we have plotted Ohmic conductivity for $e = 10$ and $e = 20$ , respectively. As it is clear from these plots Ohmic conductivity starts from a maximum value and by increasing $b$ it decreases. The main effect of increasing 't Hooft coupling constant is to decrease Ohmic conductivity value. The right plot of Fig 2 shows the same results. The point is that increasing the value of $e$ causes a decreasing of Ohmic conductivity value.

In following two paragraphs we study Hall conductivity versus $e$ and $b$ . Hall conductivity in terms of $e$ is plotted in Fig. 3 at constant $b$ . In the leftFigure 2: $\sigma_{xx}$ versus $b$ for different values of $k$ at fixed $e$ . Left: $e = 10$ . Right: $e = 20$ .

plot of this figure $b = 10$ . It is clearly seen that Hall conductivity also starts from its maximum value and it decreases by increasing $e$ . Moreover if 't Hooft coupling constant increases, the maximum value of Hall conductivity will decrease. Comparing with the left plot of Fig. 3, in the right plot Hall conductivity has a smaller value. This fact, which Hall conductivity decreases by increasing $b$ , is consistent with (22c).

Hall conductivity versus $b$ is plotted in Fig. 4 at constant $e$ . Two cases, which are $e = 10$ and $e = 20$ , are considered. As it is obviously seen, similar to Fig. 2 and 3, there is a maximum value for Hall conductivity. By increasing 't Hooft coupling constant this maximum value decreases and in fact this is the most important effect of 't Hooft coupling correction on the Hall conductivity. The right plot of Fig. 4 indicates that Hall conductivity has a smaller value when $e = 20$ .

4 $\mathcal{R}^2$ corrections to AdS-Schwarzschild black brane

We consider the curvature-squared corrections on the AdS black brane solution and study DC conductivity in this background. $\mathcal{R}^2$ corrections haveFigure 3: $\sigma_{xy}$ versus $e$ for different values of $k$ at fixed $b$ . Left: $b = 10$ . Right: $b = 30$ .

been introduced in [16, 17]. It is important to point out that the first higher derivative correction in weakly curved type IIb backgrounds enters at order $\mathcal{R}^4$ , and not $\mathcal{R}^2$ , so we will not predict effect of curvature-squared corrections on the $\mathcal{N} = 4$ SU(N) SYM. At first we consider the general $\mathcal{R}^2$ corrections in (23) and calculate Ohmic conductivity and then extend the calculation to the case of Gauss-Bonnet (GB) gravity. Fortunately, we find analytic results in both cases. Hall conductivity in the presence of curvature-squared corrections can be studied, too. Here we only discuss Ohmic conductivity.

The black brane solution of $AdS_5$ space with the curvature-squared corrections is [18]

$$d{s}^2=-\kappa \left(\frac{u^2}{R^2}\right)f(u)d{t}^2+\left(\frac{u^2}{R^2}\right)d{\vec{x}}^2+\frac{1}{\left(\frac{u^2}{R^2}\right)f(u)}d{u}^2,(23)ds^2\; =\; -\backslash kappa\backslash left(\backslash frac\{u^2\}\{R^2\}\backslash right)f(u)dt^2\; +\; \backslash left(\backslash frac\{u^2\}\{R^2\}\backslash right)d\backslash vec\{x\}^2\; +\; \backslash frac\{1\}\{\backslash left(\backslash frac\{u^2\}\{R^2\}\backslash right)f(u)\}du^2,\; \backslash quad\; (23)$$

where

$$f(u)=1-\frac{u_0^4}{u^4}+\alpha +\gamma \frac{u_0^8}{u^8}\mathrm{.}(24)f(u)\; =\; 1\; -\; \backslash frac\{u\_0^4\}\{u^4\}\; +\; \backslash alpha\; +\; \backslash gamma\; \backslash frac\{u\_0^8\}\{u^8\}.\; \backslash quad\; (24)$$

and $\alpha$ and $\gamma$ are small variables. The scaling factor $\kappa = \frac{1}{1+\alpha}$ was included for the speed of light in the boundary to be unity. Also $u$ denotes the radial coordinate of the black brane geometry and $t, \vec{x}$ label the directions along the boundary at the spatial infinity. In these coordinates the event horizonFigure 4: $\sigma_{xy}$ versus $b$ for different values of $k$ at fixed $e$ . Left: $e = 10$ . Right: $e = 20$ .

is located at $f(u_0) = 0$ where $u_0$ can be found by solving this equation. The boundary is located at infinity and the geometry will be asymptotically AdS with a radius of curvature $R = 1$ . The temperature is given by

$$T_{{\mathcal{R}}^2}=\frac{u_0}{\pi }(1+\frac{1}{4}\alpha -\frac{5}{4}\gamma )\mathrm{.}(25)T\_\{\backslash mathcal\{R\}^2\}\; =\; \backslash frac\{u\_0\}\{\backslash pi\}\; \backslash left(\; 1\; +\; \backslash frac\{1\}\{4\}\backslash alpha\; -\; \backslash frac\{5\}\{4\}\backslash gamma\; \backslash right).\; \backslash quad\; (25)$$

As what it was done in section 3.1, (8a) after setting to zero, becomes

$$w((1+\alpha )w+\frac{e^2}{\kappa }{(1+\frac{\alpha }{4}-\frac{5\gamma }{4})}^4-1)+\gamma =0,(26)w\; \backslash left(\; (1\; +\; \backslash alpha)w\; +\; \backslash frac\{e^2\}\{\backslash kappa\}\; \backslash left(\; 1\; +\; \backslash frac\{\backslash alpha\}\{4\}\; -\; \backslash frac\{5\backslash gamma\}\{4\}\; \backslash right)^4\; -\; 1\; \backslash right)\; +\; \backslash gamma\; =\; 0,\; \backslash quad\; (26)$$

where

$$e=\frac{E}{\frac{\pi }{2}\sqrt{\lambda }{T}_{{\mathcal{R}}^2}^2}\mathrm{.}(27)e\; =\; \backslash frac\{E\}\{\backslash frac\{\backslash pi\}\{2\}\backslash sqrt\{\backslash lambda\}T\_\{\backslash mathcal\{R\}^2\}^2\}.\; \backslash quad\; (27)$$

Obviously by setting $\alpha$ and $\gamma$ to zero one must find Ohmic conductivity in AdS-Schwarzschild background brought in (21). This virtue selects an acceptable root of (26) which was already called $w_*$ . It is then straightforwardto find Ohmic conductivity from (18) that is given by

where

$$\begin{array}{cccc}& M(\alpha ,\gamma ,e)=-2^{18}\gamma (1+\alpha )+(256+(1+\alpha )(4+\alpha -5\gamma {)}^4{e}^2{)}^2,& & \text{(29)}\end{array}M(\backslash alpha,\; \backslash gamma,\; e)\; =\; -2^\{18\}\; \backslash gamma(1+\backslash alpha)\; +\; (256+(1+\backslash alpha)(4+\backslash alpha-5\backslash gamma)^4\; e^2)^2,\; \backslash tag\{29\}$$

and

$$\begin{array}{cccc}& q=\frac{Q}{\frac{\pi }{2}\sqrt{\lambda }{T}_{{\mathcal{R}}^2}^2}\mathrm{.}& & \text{(30)}\end{array}q\; =\; \backslash frac\{Q\}\{\backslash frac\{\backslash pi\}\{2\}\; \backslash sqrt\{\backslash lambda\}\; T\_\{\backslash mathcal\{R\}^2\}^2\}.\; \backslash tag\{30\}$$

Regarding to small values of $\alpha$ and $\gamma$ , as it is expected, the above Ohmic conductivity reproduces (21) for large value of electric field at fixed temperature. Moreover, as original case introduced in [4], although two types of charge carries contribute to the conductivity, which are charge carries represented by $q$ and charge carries thermally produced, the value of them are corrected by $\mathcal{R}^2$ correction. For example as it was pointed out in (12), in the case of massive charge carriers $\hat{\sigma}$ dominates in (28). Based on the small values of $\alpha$ and $\gamma$ , we expand this term and keep only first order terms as

$$\begin{array}{cccc}& ({\widehat{\sigma }}_{{\mathcal{R}}^2}{)}^2=(\widehat{\sigma }{)}^2(1+\left(\frac{1-e^2}{1+e^2}\right)\alpha +\frac{1+5e^2+5e^4}{(1+e^2{)}^2}\gamma ),& & \text{(31)}\end{array}(\backslash hat\{\backslash sigma\}\_\{\backslash mathcal\{R\}^2\})^2\; =\; (\backslash hat\{\backslash sigma\})^2\; \backslash left(\; 1\; +\; \backslash left(\; \backslash frac\{1-e^2\}\{1+e^2\}\; \backslash right)\; \backslash alpha\; +\; \backslash frac\{1+5e^2+5e^4\}\{(1+e^2)^2\}\; \backslash gamma\; \backslash right),\; \backslash tag\{31\}$$

where

$$\begin{array}{cccc}& (\widehat{\sigma }{)}^2=\frac{q}{1+e^2}\mathrm{.}& & \text{(32)}\end{array}(\backslash hat\{\backslash sigma\})^2\; =\; \backslash frac\{q\}\{1+e^2\}.\; \backslash tag\{32\}$$

In five dimensions, the most general theory of gravity with quadratic powers of curvature is GB theory. The exact solutions and thermodynamic properties of the black brane in GB gravity were discussed in [19, 20, 21]. We are going to more understand about the DC conductivity in the GB gravity. The black brane solution in this geometry is given by [19]

$$\begin{array}{cccc}& d{s}^2=-a\frac{u^2}{R^2}h(u)d{t}^2+\frac{d{u}^2}{\frac{u^2}{R^2}h(u)}+\frac{u^2}{R^2}d{\vec{x}}^2,& & \text{(33)}\end{array}ds^2\; =\; -a\; \backslash frac\{u^2\}\{R^2\}\; h(u)\; dt^2\; +\; \backslash frac\{du^2\}\{\backslash frac\{u^2\}\{R^2\}\; h(u)\}\; +\; \backslash frac\{u^2\}\{R^2\}\; d\backslash vec\{x\}^2,\; \backslash tag\{33\}$$where

$$h(u)=\frac{1}{2{\lambda }_{GB}}[1-\sqrt{1-4{\lambda }_{GB}(1-\frac{u_0^4}{u^4})}]\mathrm{.}(34)h(u)\; =\; \backslash frac\{1\}\{2\backslash lambda\_\{GB\}\}\; \backslash left[\; 1\; -\; \backslash sqrt\{1\; -\; 4\backslash lambda\_\{GB\}\; \backslash left(\; 1\; -\; \backslash frac\{u\_0^4\}\{u^4\}\; \backslash right)\}\; \backslash right].\; \backslash quad\; (34)$$

In (33), $a$ is an arbitrary constant which specifies the speed of light of the boundary gauge theory and we choose it to be unity. As a result at the boundary, where $u \rightarrow \infty$ ,

$$h(u)\to \frac{1}{a},a=\frac{1}{2}(1+\sqrt{1-4{\lambda }_{GB}})\mathrm{.}(35)h(u)\; \backslash rightarrow\; \backslash frac\{1\}\{a\},\; \backslash quad\; a\; =\; \backslash frac\{1\}\{2\}\; \backslash left(\; 1\; +\; \backslash sqrt\{1\; -\; 4\backslash lambda\_\{GB\}\}\; \backslash right).\; \backslash quad\; (35)$$

We assume $\lambda_{GB} \leq \frac{1}{4}$ , the reason is that beyond this point there is no vacuum AdS solution and one cannot have a conformal field theory at the boundary. The temperature is given by

$$T_{GB}=\frac{\sqrt{a}{u}_0}{\pi }\mathrm{.}(36)T\_\{GB\}\; =\; \backslash frac\{\backslash sqrt\{a\}\; u\_0\}\{\backslash pi\}.\; \backslash quad\; (36)$$

In this case (8a) and (18) lead to

$$w^4(1-\sqrt{1-4{\lambda }_{GB}(1-\frac{1}{w})})-2a{e}^2{\lambda }_{GB}=0,(37)w^4\; \backslash left(\; 1\; -\; \backslash sqrt\{1\; -\; 4\backslash lambda\_\{GB\}\; \backslash left(\; 1\; -\; \backslash frac\{1\}\{w\}\; \backslash right)\}\; \backslash right)\; -\; 2ae^2\; \backslash lambda\_\{GB\}\; =\; 0,\; \backslash quad\; (37)$$

and

where

$$g({\lambda }_{GB},e)=2(1+2a{e}^2)+2e^4(a-{\lambda }_{GB})(1+{\lambda }_{GB}),(39)g(\backslash lambda\_\{GB\},\; e)\; =\; 2(1+2ae^2)\; +\; 2e^4(a-\backslash lambda\_\{GB\})(1+\backslash lambda\_\{GB\}),\; \backslash quad\; (39)$$

and

$$e=\frac{E}{\frac{\pi }{2}\sqrt{\lambda }{T}_{GB}^2},q=\frac{Q}{\frac{\pi }{2}\sqrt{\lambda }{T}_{GB}^2}\mathrm{.}(40)e\; =\; \backslash frac\{E\}\{\backslash frac\{\backslash pi\}\{2\}\backslash sqrt\{\backslash lambda\}\; T\_\{GB\}^2\},\; \backslash quad\; q\; =\; \backslash frac\{Q\}\{\backslash frac\{\backslash pi\}\{2\}\backslash sqrt\{\backslash lambda\}\; T\_\{GB\}^2\}.\; \backslash quad\; (40)$$

It is clearly seen that by setting $\lambda_{GB} = 0$ , one finds the Ohmic conductivity in AdS-Schwarzschild background. Interpretation of two terms contributing to Ohmic conductivity in (38) is the same as $\mathcal{R}^2$ correction case.## 5 Discussion and Conclusion

In this paper effect of curvature correction on DC conductivity is studied. In particular we considered $\mathcal{R}^4$ correction to AdS-Schwarzschild black brane. Our results show that there is a critical value for electric field in which correction to Ohmic conductivity vanishes. Moreover it was shown that, depending on other parameters, Ohmic conductivity can increase or decrease. In another case, when magnetic field is turned on, Hall and Ohmic conductivities are plotted in Fig. 1-4. At fixed temperature and large magnetic field, Ohmic and Hall conductivity generally start from their maximum value. Fig. 4 shows that Hall conductivity has a maximum value at fixed electric field and temperature.

Curvature-squared and Gauss-Bonnet corrections are then considered in the next section. As it is expected, the main structure of Ohmic conductivity is preserved by corrections.

It is straightforward to calculate the DC conductivity from the drag force calculations. One should consider massive carriers as endpoint of strings which end on flavor branes and using the quasi-particle description write the equation of motion for them at the equilibrium where the external force is $f = E$ . At large mass limit, only charge carriers contribute to current and one may express $\langle J^x \rangle$ in terms of velocity of the quasi-particles, $\langle J^x \rangle = \langle J^t \rangle v$ . Regarding Ohm's law, we have $v = \frac{\sigma E}{\langle J^t \rangle}$ , where $v$ is velocity of massive carrier and it is constant. One can follow this approach and derive $\hat{\sigma}$ in the case of $\mathcal{R}^2$ and Gauss-Bonnet corrections in (28) and (38). This approach has been followed in the case of strange metals in [7, 8].

Acknowledgment

M. A. would like to thank M. M. sheikh-Jabbari for instructive discussions. We thank the organizers of ISS2010 for providing an excellent atmosphere for physics discussions. We would like to thank Carlos Nunez for valuable discussions and comments.

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