Field-Angle Dependence of Interlayer Magnetoresistance in Organic Dirac Electron System α-(BEDT-TTF)₂I₃

Abstract

The effect of the Coulomb interaction in interlayer magnetoresistance is elucidated in collaboration with theory and experiments for the Dirac electron system in organic conductor $\alpha$-(BEDT-TTF)${}_2$I${}_3$ under a strong magnetic field. It is found that the effective g-factor enhanced by Coulomb interaction depends on the angle of the magnetic field, resulting in the field-angle dependence of a characteristic magnetic field in which interlayer resistance has a minimum due to spin splitting $N=0$ Landau levels. The qualitative agreement between the theory and experimental results for the field-angle dependence of interlayer magnetoresistance is obtained.

1. Introduction

The electron correlation effects in two-dimensional Dirac electron systems have attracted much attention [1,2,3,4,5]. In the Dirac electron system of organic conductor $\alpha$-(BEDT-TTF)${}_2$I${}_3$ [6,7,8,9,10,11,12,13], it was shown that the electron correlation effects become a key factor to understanding electronic properties [14,15,16,17,18,19,20,21,22], since the Coulomb interaction is comparable with the band width. Moreover, the Fermi energy almost coincides with the Dirac point in $\alpha$-(BEDT-TTF)${}_2$I${}_3$; thus, any other energy bands do not overlap with Fermi energy [23,24]. $\alpha$-(BEDT-TTF)${}_2$I${}_3$ has a clean Dirac electron system, since the density of impurity is estimated to the ppm order [23,24]. These features are also advantageous to developing the physics of the correlated Dirac electron system.

The layered structure of $\alpha$-(BEDT-TTF)${}_2$I${}_3$ enables interlayer magnetoresistance measurements, which revealed the anomalous electronic properties of two-dimensional Dirac electron systems connected by weak interlayer tunneling [25,26,27,28,29,30]. In the magnetic field normal to the conductive layer, the energy of Landau levels in a massless Dirac electron system is expressed as $E_N=\pm \sqrt{2e\hslash v_{\mathrm{F}}^2\left|N\right|B}$, where ℏ, $v_{\mathrm{F}}$, N, and B denote the Planck constant, the Fermi velocity of the Dirac cone, the Landau index, and the magnetic-field strength, respectively. One of the characteristic features in these systems is the appearance of $N=0$ Landau levels at the Dirac points. This effect was detected in interlayer magnetoresistance under a transverse magnetic field [25,26]. Interlayer magnetoresistance primarily depends on the interlayer tunneling of the Landau carriers, where Landau carriers indicate the carriers belonging to Landau levels that contribute to electric current. Note that in each Landau levels there are states with density proportional to B. Thus, the magnetic field creates mobile N = 0 Landau level carriers. The effect of the magnetic field appears only through the change of the N = 0 Landau level carrier density at the vicinity of the Dirac points. Thus, negative interlayer magnetoresistance due to the increase of the degeneracy of the $N=0$ Landau levels was observed [25,26]. It was also shown that interlayer resistance has a minimum for $g{\mu }_{\mathrm{B}}{B}_0/2\cong \hslash /\tilde{\tau }$ due to the Zeeman splitting of the $N=0$ Landau levels, where g, ${\mu }_{\mathrm{B}}$, and $\tilde{\tau }$ denote the g-factor, the Bohr magneton, and the relaxation time, respectively. If the electron correlation effects in the Landau levels are negligible, $B_0$ is independent of the angle of the magnetic field.

The electron correlation effects in the Landau levels, however, have been controversial. Although the possible ordered states due to Coulomb interaction, such as the valley-ordered state [31,32,33] and the interlayer spin-ordered state [34,35], were proposed, it was suggested that the anomalous increase of the spin lattice relaxation rate at low temperatures [33] can be explained by the spin transverse fluctuation in the absence of ordered states [36].

In the present study, we investigate the effects of the electron correlation between N = 0 Landau level carriers on interlayer magnetoresistance as a function of field-angle $\theta$ from the interlayer axis in collaboration with theory and experiment. The effective g-factor, $g^{*}$, is treated using the mean field theory of the Coulomb interaction between the tilted Dirac electrons in the quantum limit. It is numerically shown that effective Coulomb interaction $V_{\mathrm{HS}}$, which enhances $g^{*}$, is approximately proportional to ${(Bcos\theta )}^{\gamma }$, where $\gamma$ depends on the tilt of the Dirac cone. It is found that a characteristic magnetic field $B_0$, at which the interlayer resistance has a minimum, depends on $\theta$ and temperature T, where the inverse of $B_0$ is proportional to $cos\theta$ approximately and the coefficient increases as T decreases. These results are in qualitative agreement with the experiment.

2. Method

2.1. Formulation

In $\alpha$-(BEDT-TTF)${}_2$I${}_3$, there are two band-crossing points called Dirac points being assigned as the right (R) and left (L) valleys. The effective Hamiltonian describing the Dirac electron system in $\alpha$-(BEDT-TTF)${}_2$I${}_3$ is given by [10,31]

$$H=H_0+H^{\prime },$$

(1)

where kinetic energy term $H_0$ is

$$\begin{array}{c}\hfill H_0=\sum _{\mathbf{q}\gamma {\gamma }^{\prime }\tau s}{a}_{\mathbf{r}\gamma ,\tau s}^{†}{[{\widehat{H}}_0^{\tau s}]}_{\gamma {\gamma }^{\prime }}{a}_{\mathbf{r}{\gamma }^{\prime },\tau s},\end{array}$$

(2)

$$\begin{array}{c}\hfill {\widehat{H}}_0^{\tau s}=-\mathrm{i}\tau \hslash v\left(\begin{array}{cc}\eta {\partial }_x& {\partial }_x-\mathrm{i}\tau \partial {}_y\\ {\partial }_x+\mathrm{i}\tau {\partial }_y& \eta {\partial }_x\end{array}\right),\end{array}$$

(3)

where $a_{\mathbf{r}\gamma ,\tau s}^{†}$ and $a_{\mathbf{r}\gamma ,\tau s}$ represent creation and annihilation operators, respectively, with two dimensional space $\mathbf{r}=(x,y)$, Luttinger–Kohn base $\gamma$ [10,37], valley $\tau =\pm$ (R, L), and spin $s=\pm$ (↑, ↓). The degree of tilt $\eta$ is defined by $\eta =v_0/v$ with cone velocity v and tilt velocity $v_0$, where the anisotropy of the cone velocity is ignored here for simplicity [31]. The energy eigenvalue of $H_0$ is given by

$$E=\hslash v\left(\eta k_x\pm \sqrt{k_x^2+k_y^2}\right),$$

(4)

with two-dimensional momentum $k_x$ and $k_y$. The left inset in Figure 1 shows the tilted Dirac cone, where $v\pm v_0$ are velocities in the $\pm k_x$ directions, respectively. Interaction term ${\widehat{H}}^{\prime }$ is given by

$${\widehat{H}}^{\prime }=\frac{1}{2}\int \mathrm{d}\mathbf{r}\int \mathrm{d}{\mathbf{r}}^{\prime }V(\mathbf{r}-{\mathbf{r}}^{\prime })n(\mathbf{r})n({\mathbf{r}}^{\prime })$$

(5)

with long-range Coulomb interaction $V(\mathbf{r})=e^2/\epsilon r$ and electron density operator $n(\mathbf{r})$.

The energy spectrum of the two-dimensional electronic system is quantized under a tilted magnetic field, $\mathbf{B}=\nabla \times \mathbf{A}=(B_x,B_y,B_z)$, given by the vector potential with the Landau gauge, $\mathbf{A}=(B_{y}z-B_{z}y,-B_{x}z,0)$. The Hamiltonian under the magnetic field is obtained by Peierls substitution $-i\nabla \to -i\nabla +(e/\hslash )\mathbf{A}$ and Zeeman energy $E_{\mathrm{Z}}=g{\mu }_{\mathrm{B}}B/2$ with $B=\left|\mathbf{B}\right|$. The Landau levels are given by $E_{Ns}=\mathrm{sgn}(N)(\hslash v/l)\sqrt{2{\lambda }^3\left|N\right|}-s{E}_{\mathrm{Z}}$ with $\lambda =\sqrt{1-{\eta }^2}$ and magnetic length $l=\sqrt{\hslash /e|B_z|}$. The wave function ${\mathsf{\Psi }}_{N,k}^{\tau }(\mathbf{r})$ for the $N=0$ Landau level is given by References [11,27,38]

$$\begin{array}{ccc}\hfill & & {\mathsf{\Psi }}_{N=0,k}^{\tau =+}(\mathbf{r})=\frac{1}{\sqrt{2(1+\lambda )}}\left(\begin{array}{c}-\eta \\ 1+\lambda \end{array}\right){\varphi }_{N=0,k}(\mathbf{r}),\hfill \end{array}$$

(6)

$$\begin{array}{cc}& {\mathsf{\Psi }}_{N=0,k}^{\tau =-}(\mathbf{r})=\frac{1}{\sqrt{2(1+\lambda )}}\left(\begin{array}{c}-1-\lambda \\ \eta \end{array}\right){\varphi }_{N=0,k}(\mathbf{r}),\hfill \end{array}$$

(7)

where

$${\varphi }_{N=0,k}(\mathbf{r})=\frac{{\lambda }^{1/4}}{\sqrt{2\pi }}\frac{1}{{\left(\sqrt{\pi }l\right)}^{1/2}}{e}^{ikx}{e}^{-{\tilde{Y}}^2/2}$$

(8)

with $\tilde{Y}=\frac{\sqrt{\lambda }}{l}(y-Y)$ and center coordinate $Y=l^{2}k$. When $H=5$ T, $E_1\cong 3.5$ meV using values of parameters for $\alpha$-(BEDT-TTF)${}_2$I${}_3$, where velocity $v=1.0\times {10}^5$ m/s and $v_0=0.8\times {10}^5$ m/s are given by the band calculation [10,23,31], $2E_{\mathrm{Z}}\cong 0.5$ meV with $g=2$, $l\cong 14$ nm.

In the present study, we consider the $N=0$ Landau levels in order to study interlayer magnetoresistivity in the quantum limit and, for the case of $E_1\gg E_{\mathrm{Z}}$. The effective g-factor, $g^{*}$, is treated by the mean field theory. The Green function $G_s(k,\mathrm{i}{\epsilon }_n)$ is defined by

$$G_s(k,\mathrm{i}{\epsilon }_n)=\frac{1}{\mathrm{i}{\epsilon }_n+\mu +s{E}_{\mathrm{Z}}-{\mathsf{\Sigma }}_s},$$

(9)

where ${ϵ}_n=(2n+1)\pi /\beta$ is fermion Matsubara frequency with $\beta =1/k_{\mathrm{B}}T$ and integer n, and $\mu$ is the chemical potential, determined so that the Fermi energy coincides with the Dirac point. The self-energy ${\mathsf{\Sigma }}_s$ is given by self-consistent equation

$${\mathsf{\Sigma }}_{\uparrow }-{\mathsf{\Sigma }}_{\downarrow }=-V_{\mathrm{HS}}{m}_z,$$

(10)

with effective Coulomb interaction $V_{\mathrm{HS}}={\sum }_{{\tau }^{\prime }}{[V(0)]}_{\tau ,\tau ,{\tau }^{\prime },{\tau }^{\prime }}$, magnetization $m_z=n_{\uparrow }-n_{\downarrow }$, and electron density for spin s, $n_s$, where

$${\displaystyle {\mathsf{\Sigma }}_s=\frac{1}{D}\sum _{k^{\prime }}\frac{1}{\beta }\sum _{{\epsilon }_n^{\prime }}\sum _{{\tau }^{\prime }}{[V(0)]}_{\tau ,\tau ,{\tau }^{\prime },{\tau }^{\prime }}{G}_{-s}(k^{\prime },\mathrm{i}{\epsilon }_n^{\prime })}$$

(11)

and the Coulomb interaction matrix ${[V(q)]}_{{\tau }_1{\tau }_2,{\tau }_3,{\tau }_4}$ for the $N=0$ Landau levels is given by

$$\begin{array}{cc}\hfill & {[V(q)]}_{{\tau }_1{\tau }_2,{\tau }_3,{\tau }_4}=\frac{1}{2}\int \mathrm{d}\mathbf{r}\int \mathrm{d}{\mathbf{r}}^{\prime }V(\mathbf{r}-{\mathbf{r}}^{\prime })\times \hfill \\ \hfill & [{\mathsf{\Psi }}_{N=0,k+q}^{{\tau }_2}{(\mathbf{r})}^{†}·{\mathsf{\Psi }}_{N=0,k}^{{\tau }_1}(\mathbf{r})][{\mathsf{\Psi }}_{N=0,k^{\prime }-q}^{{\tau }_4}{({\mathbf{r}}^{\prime })}^{†}·{\mathsf{\Psi }}_{N=0,k^{\prime }}^{{\tau }_3}({\mathbf{r}}^{\prime })],\hfill \end{array}$$

(12)

where the degeneracy of center coordinate $D=L_x{L}_y/2\pi l^2$ with length $L_x$ and $L_y$ in the x and y directions, respectively. The effective Coulomb interaction depends on magnetic length l, so effective Coulomb interaction depends on angle $\theta$. Effective spin splitting $E_{\mathrm{Z}}^{*}$ is given by

$$E_{\mathrm{Z}}^{*}=g^{*}{\mu }_{\mathrm{B}}B/2=E_{\mathrm{Z}}+\mathsf{\Delta }$$

(13)

with $\mathsf{\Delta }={\mathsf{\Sigma }}_{\downarrow }=-{\mathsf{\Sigma }}_{\uparrow }\ge 0$ for the charge neutral system $\mu =0$. Thus, effective g-factor $g^{*}$ is given by

$$g^{*}=g+2\mathsf{\Delta }/{\mu }_{\mathrm{B}}B.$$

(14)

Thus, the energy eigenvalues of N = 0 Landau levels are modified as follows:

$$E_{N=0,s}=-s{E}_Z^{*}=-s(E_Z+\mathsf{\Delta }).$$

(15)

Interlayer conductivity is given by interlayer coupling as a perturbation [25]. The perturbation Hamiltonian $H^{\prime }$ is given by

$${\widehat{H}}^{\prime }=-2t_{c}cos\left(-ic\frac{\partial }{\partial z}\right)\left(\begin{array}{cc}1& 0\\ 0& 1\end{array}\right)$$

(16)

where $t_c$ and c represent interlayer transfer energy and interlayer spacing, respectively. In the quantum limit, N = 0 Landau levels are dominant in magnetotransport. The effective transfer energy between N = 0 Landau levels in neighboring layers is given by [25]:

$$\begin{array}{ccc}\hfill \widetilde{t_c}(Y^{\prime },z_i^{\prime };Y,z_i)& =& t_c\times exp\left[-\frac{1}{4}\frac{c^{2}e\left(B_x^2+B_y^2\right)}{\hslash |B_z|}\right]\hfill \\ & & \times exp\left[i\frac{e{B}_x}{\hslash }(z_i^{\prime }-z_i)\frac{Y+Y^{\prime }}{2}\right],\hfill \end{array}$$

(17)

where $z_i$ is the layer position, and the neighboring layers are $z_i^{\prime }=z_i\pm c$. The center coordinate of initial state Y on one layer $z=z_i$, and that of final state $Y^{\prime }$ on neighboring layer $z=z_i\pm c$ satisfy the condition

$$Y^{\prime }=Y\pm \frac{B_y}{B_z}c.$$

(18)

The complex interlayer conductivity ${\tilde{\sigma }}_{zz}(\omega )$ is given by [25]:

$$\begin{array}{ccc}\hfill {\tilde{\sigma }}_{zz}(\omega )=-\frac{i\hslash }{L^2}& {\displaystyle \sum _{Y,z_i,\tau ,s;Y^{\prime },z_i^{\prime },{\tau }^{\prime },s^{\prime }}}& \langle N=0,Y,z_i,\tau ,s\left|{\widehat{j}}_z\right|N=0,Y^{\prime },z_i^{\prime },{\tau }^{\prime },s^{\prime }\rangle \hfill \\ & & \times \langle N=0,Y^{\prime },z_i^{\prime },{\tau }^{\prime },s^{\prime }\left|{\widehat{j}}_z\right|N=0,Y,z_i,\tau ,s\rangle \hfill \\ & & \times \frac{f(E_{N=0,s})-f(E_{N=0,s^{\prime }})}{E_{N=0,s^{\prime }}-E_{N=0,s}}\frac{1}{E_{N=0,s^{\prime }}-E_{N=0,s}-\hslash \omega -i\hslash /\tilde{\tau }},\hfill \end{array}$$

(19)

where $\tilde{\tau }$ and ${\widehat{j}}_z$ represent relaxation time and interlayer current density, respectively. The center coordinate Y is associated with wavenumber k by relation expression $Y=l^{2}k$. Interlayer current density is given by ${\widehat{j}}_z=(-e)(1/i\hslash )[\widehat{z},{\widehat{H}}^{\prime }]$.

The leading term of real conductivity is given by [25]:

$${\sigma }_{zz}=\frac{2C{t}_c^{2}c{e}^3\tilde{\tau }\left|B_z\right|}{\pi {\hslash }^3}exp\left[-\frac{e{c}^2(B_x^2+B_y^2)}{2\hslash |B_z|}\right]$$

(20)

with

$$C=\sum _{s\tau }\int D_{s\tau }{(E)}^2\left(-\frac{\mathrm{d}f}{\mathrm{d}E}\right)\mathrm{d}E$$

(21)

where $D_{s\tau }(E)$, $t_c$ and c denote density of states for spin s and valley $\tau$, interlayer transfer energy, and interlayer spacing, respectively. Interlayer resistivity ${\rho }_{zz}$ is given by ${\rho }_{zz}\simeq 1/{\sigma }_{zz}$, since interlayer Hall conductivities ${\sigma }_{xz}$ and ${\sigma }_{yz}$ are negligibly smaller than other components [39,40].

2.2. Experimental Method

2.2.1. Crystal Growth

Either the electrolysis method or the diffusion method are generally used in the crystal growth of organic conductors. We synthesized organic conductor $\alpha$-(BEDT-TTF)${}_2$I${}_3$ by the electrolysis method using an H-type cell. BEDT-TTF molecules and I${}_3^{-}$ anions are desolved in a supporting electrolyte (THF, benzonitrile, chlorobenzene, etc.). Then, we supply electrical current (1∼5 $\mathsf{\mu }$A) between platinum electrodes. After about 1∼2 weeks, small single crystals appear on the positively based platinum electrode. The typical size of a crystal is $1\times 0.5\times 0.05$ mm${}^3$.

2.2.2. Experiments of Interlayer Magnetoresistance Under Pressure

A sample with a dimension of approximately 0.7 × 0.5 × 0.05 mm${}^3$, on which four electrical leads (gold wire with a diameter of 15 $\mathsf{\mu }$m) are attached by carbon paste, is put in a Teflon capsule filled with the pressure medium (Idemitsu DN-oil 7373); then, the capsule is set in a NiCrAl clamp cell, and hydrostatic pressure of up to 1.7 GPa is applied. The hydrostatic pressure is determined at room temperature by a Manganine resistance gauge in the pressure cell. The interlayer resistance of a crystal is measured by a conventional DC method with an electrical current of 1 $\mathsf{\mu }$A along the c-crystal axis, which is normal to the two-dimensional plane. In the investigation, interlayer magnetoresistance is measured as functions of B and $\theta$ which is the angle between the magnetic-field direction and c-crystal axis at $T=$ 0.5, 1.7, 2.5, 3.0, 3.5, and 4.2 K. As mentioned in the introduction, interlayer magnetoresistance is a useful tool to detect the effects of N = 0 Landau levels, including its Zeeman splittings.

3. Results

Figure 1 shows the theoretical results on $|Bcos\theta |$ ($=|B_z|$) dependences of effective Coulomb interaction $V_{\mathrm{HS}}$ for tilt parameter $\eta =0$, $0.5$, $0.8$, and $0.9$. It is numerically shown that $V_{\mathrm{HS}}\propto {|Bcos\theta |}^{\gamma }$ approximately for $|Bcos\theta |>3$. Effective Coulomb interaction depends on magnetic length l, which is a function of $|B_z|$, as shown in Equation (12). Thus, effective Coulomb interaction depends on angle $\theta$. The left inset shows the tilting Dirac cone, where v and $v_0$ represent cone velocity and tilt velocity, respectively. The right inset shows the $\eta$ dependence of $\gamma$, where $\gamma$ increases as $\eta$ increases. Thus, we use a relation, $V_{\mathrm{HS}}=u{|Bcos\theta |}^{\gamma }$, with $\gamma =0.87$ for the tilted Dirac cones in $\alpha$-(BEDT-TTF)${}_2$I${}_3$ with $\eta =0.8$ [23] hereafter. Parameter $u=0.3$ is chosen to fit with the experimental results.

Figure 2a,b shows the theoretical results on the B-dependences of $g^{*}$ and $E_{\mathrm{Z}}^{*}$, respectively, for $\theta =0$, 20, 40, and ${60}^{\circ }$ at $T=1.7$ K. It is found that both $g^{*}$ and $E_{\mathrm{Z}}^{*}$ enhance by $V_{\mathrm{HS}}$ depend on $\theta$. When $\theta ={90}^{\circ }$, $g^{*}=g$ and $E_{\mathrm{Z}}^{*}=E_{\mathrm{Z}}$, since $V_{\mathrm{HS}}=0$. Although $E_{\mathrm{Z}}^{*}$ increases monotonically as B increases, $g^{*}$ has a maximum since $\mathsf{\Delta }$ divided by B contributes to $g^{*}$.

Figure 3a shows the theoretical results on B-dependences of interlayer resistivity ${\rho }_{zz}$ for $\theta =0$, 20, 40, and ${60}^{\circ }$ at $T=1.7$ K. ${\rho }_{zz}$ has a minimum at $B_0$. It is found that $B_0$ increases as $\theta$ increases due to $\theta$-dependence of $E_{\mathrm{Z}}^{*}$. Figure 3b shows the experimental results on B-dependences of interlayer resistance $R_{zz}$ for $\theta =0$, 20, 40, and ${60}^{\circ }$ at $T=1.7$ K. $B_0$ obtained in the experimental results also increases as $\theta$ increases.

In a general two-dimensional system, $E_{\mathrm{Z}}^{*}$ dose not depend on $\theta$. The agreement between the theory and experiment of interlayer magnetoresistance shown in Figure 3 indicates that effective Coulomb interaction plays an important role to the Zeeman effects. In the following, peculiar Zeeman effects in this system are examined.

The first step is to investigate $g^{*}$ for $\theta$ = 0 from the interlayer-magnetoresistance minimum, where $g^{*}{\mu }_{\mathrm{B}}{B}_0\sim 2\hslash /\tilde{\tau }$. Here, the rough of broadening energy $\hslash /\tilde{\tau }$ of the Landau levels in this system is 3 K at low temperatures [32]. $g^{*}$ for $\theta =0$ is roughly estimated to be 5 experimentally at 1.7 K; this is close to the theoretical value, which is approximately 5.3 at $B_0\sim 1.8$ T, as shown in Figure 2a.

Lastly, the peculiar Zeeman effects on the $\theta$-dependence of the interlayer magnetoresistance minimum are detected. In Figure 4a, the theoretical results on $\theta$ dependences of $B_0^{-1}$ are drawn as functions of $cos\theta$ for $T=0.5$, $1.7$, $2.5$, $3.0$, $3.5$, and $4.2$ K. It is numerically shown that $1/B_0\cong acos\theta +b$ when $\theta$ is close to $0^{\circ }$. Note that this numerical calculation is not applicable when $\theta$ is close to ${90}^{\circ }$, where contributions of higher Landau levels in interlayer resistivity are not negligible. Figure 4b shows the experimental results on $cos\theta$ dependences of $B_0^{-1}$ for $T=0.5$, $1.7$, $2.5$, $3.0$, $3.5$, and $4.2$ K. The experimental results also show the same approximate relation on $B_0^{-1}$ as a linear function of $cos\theta$.

Figure 5 shows the theoretical and experimental results on T dependencies of coefficient a. It is found that coefficient a increases as T decreases, indicating remarkable $\theta$ dependence of $B_0^{-1}$ at very low temperatures $T\le 1.7$ K. Those results show qualitative agreement between theory and experimental results for the field-angle dependence of interlayer magnetoresistance.

4. Discussion

Those theoretical curves in Figure 3a and Figure 4a qualitatively reproduce the experimental results including the characteristic features of the resistance minimum as shown in Figure 3b and Figure 4b. Here, the theoretical results do not coincide with the experimental results near B = 0 T, since only N = 0 Landau levels are examined in the present theoretical calculation. This theoretical approach, however, is valid because the special Landau-level structure in this system realizes the quantum limit in the magnetic field above $0.07$ T for a perpendicular component to the two-dimensional plane at $1.7$ K [32,41].

In the present study, the value of u for $V_{\mathrm{HS}}$ is chosen to fit with the experimental results. The value of u will be evaluated by taking the Thomas–Fermi screening effect into account. The effects of the Coulomb interaction in $N\ne 0$ Landau levels is also going to be studied in the mean field calculation. In addition, interlayer magnetoresistance is also going to be studied, taking $N\ne 0$ Landau levels into account, which leads to the maximum of the interlayer resistance under weak magnetic fields [26,28].

5. Conclusions

In conclusion, the effect of the Coulomb interaction in interlayer magnetoresistance was elucidated in collaboration with theory and experiments for the Dirac electron system in organic conductor $\alpha$-(BEDT-TTF)${}_2$I${}_3$. It was shown that enhancement of the effective g-factor due to the Coulomb interaction for $N=0$ Landau levels depends on field angle $\theta$. This was the key factor to explain the field-angle dependence of $B_0$ at which interlayer resistance has a minimum.

The value of the effective g-factor obtained in the present study at $\theta =0$ under a strong magnetic field is consistent with the theoretical and experimental results of the Nernst effect [42,43]. This is also consistent with the theoretical and experimental results of the spin-lattice relaxation rate [33,36]. The quantum Hall ferromagnetic state assumed in the present study supports the helical surface state [29].