Ultrafast Pump–Probe Spectroscopy in Organic Dirac Electron Candidate α-(BETS)₂I₃

Abstract

Photo-induced carrier dynamics were measured in the organic Dirac electron candidate $\alpha$-(BETS)${}_2$I${}_3$ to investigate why resistivity increases below $T_{\mathrm{MI}}$ = 50 K. We found a change in carrier dynamics due to an insulating gap formation below $T^{\prime }$ = 50 K. On the other hand, the relaxation time and polarization anisotropy of the observed dynamics differ from those in the charge-ordering (CO) state of the isostructural salt $\alpha$-(ET)${}_2$I${}_3$. Based on the difference, it can be concluded that the insulating phase has a different origin than the CO state.

1. Introduction

Organic molecular conductors have been widely studied due to their rich variety of electronic phases due to strong electron correlations [1,2]. Among them, $\alpha$-(BETS)${}_2$I${}_3$ (hereafter $\alpha$-BETS), where BETS denotes bis(ethylenedithio)tetraselenafulvalene [3,4], has attracted attention as a candidate of the Dirac electron system [5,6,7,8], which has a linear energy dispersion in the band structure at ambient pressure, expecting unique electronic properties such as temperature-independent resistivity [9,10]. On the other hand, resistivity gradually increases with a decreasing temperature below $T_{\mathrm{MI}}$ = 50 K and a step-like change at around 40 K, and these origins are still controversial [11]. To date, theoretical studies [12,13], as well as various transport and magnetic measurements [14,15,16,17,18,19], have been conducted to elucidate the rise in resistivity. However, time-resolved spectroscopic measurements are still lacking.

Pump–probe time-resolved spectroscopy using femtosecond optical pulses has often been used to study the electronic properties of strongly correlated electron systems. In time-resolved spectroscopy, even if an electron system is perturbed by light on a large energy scale, the carrier relaxation process allows us to indirectly observe the electronic state as if it were unperturbed (not excited), and to capture small energy gaps and anisotropy. In fact, in organic conductors, this method has been utilized to study correlation-induced insulating states [20,21], and has contributed to elucidating their electronic properties. Thus, by measuring the carrier dynamics in $\alpha$-BETS, we can gain new insights into the origin of the increase in resistivity at low temperatures.

In this paper, photo-induced carrier relaxation dynamics in $\alpha$-BETS are reported. The signal amplitude of the dynamics begins to increase at $T^{\prime }$ = 50 K, which agrees with $T_{\mathrm{MI}}$, indicating the formation of an energy gap. Moreover, the gap amplitude estimated from the fitting analysis almost agrees with that estimated from the resistivity measurements. On the other hand, the observed dynamics are different from that in a charge-ordering (CO) state of the isostructural salt $\alpha$-(ET)${}_2$I${}_3$ (hereafter $\alpha$-ET), where ET denotes bis(ethylenedithio)-thiotetrathiafulvalene, with respect to relaxation time and polarization anisotropy. Therefore, the origin of the resistivity increase is likely to be an insulating phase different from the CO states.

2. Materials and Methods

Single crystals of $\alpha$-BETS were synthesized electrochemically [3]. Figure 1a shows schematic illustrations of BETS and ET molecules. The crystal consists of an alternating structure of conducting layer of BETS molecules and an insulating layer of I${}_3$. As shown in Figure 1b, BETS molecules are arranged and form a conducting layer.

Figure 1c shows the schematic view of the setup for a pump–probe measurement. The measurements were made with 120 fs laser pulses centered at 1.51 eV obtained from a cavity-dumped mode-lock Ti:sapphire oscillator. A repetition rate was set as 54 kHz to avoid the heating effect. Pulses were separated into two paths; one was used for a probe, while the other was changed to pulses centered at 3.02 eV by a standard frequency doubling for a pump. The pump and probe beams were superimposed on the same axis and incident perpendicular to the conduction (ab) plane of the sample. The polarization of the probe was changed by rotating the half-wave plate, and the polarization angle was measured from a direction tilted 45 degrees from the a axis. The spot sizes of the pump and probe beams were ∼20 $\mathsf{\mu }$m and ∼12 $\mathsf{\mu }$m in diameter, respectively.

In pump–probe measurement, after excitation by the pump pulse, the carriers relax immediately and accumulate in electronic states near the Fermi energy, forming the non-equilibrium occupation of carriers as well as phonons [23]. In the subsequent probing process, the non-equilibrium carrier distribution is measured as a transient change in reflectivity ($\Delta R/R$). When a gap for a low-energy electronic excitation such as an insulating gap is formed at low temperatures, a relaxation bottleneck occurs [24,25], leading to significant changes in $\Delta R/R$, such as an increase or decrease in the signal amplitude and long relaxation. Therefore, the gap formation can be probed by measuring the temperature dependence. Moreover, by measuring probe polarization dependence, we can obtain information on the anisotropic ordering of electrons, such as the CO state [21,22]. The data were taken with increasing temperature with the pump fluence of F = 59 $\mathsf{\mu }$J/cm${}^2$.

3. Results

Figure 2a,b show the transient change of reflectivity ($\Delta R/R$) from $\theta$ = 0${}^{\circ }$, 45${}^{\circ }$ (a axis), 90${}^{\circ }$, 135${}^{\circ }$ (b axis), 180${}^{\circ }$, 225${}^{\circ }$ (a axis), 270${}^{\circ }$, 315${}^{\circ }$ (b axis), and 360${}^{\circ }$ at T = 20 K and 120 K, respectively. At T = 120 K, $\Delta R/R$ changes depend on $\theta$. When the temperature changes from 120 K to 20 K, the signal amplitude increases for all values of $\theta$. Figure 2c,d show the polar plots of the signal amplitude at T = 20 K and 120 K, respectively. At T = 120 K, the signal is enhanced in the b axis direction, the trend of which does not change at T = 20 K.

To decompose the transient data into polarization-dependent (anisotropic) and -independent (isotropic) dynamics, we tried the following analyses. Since the probe beam is linearly polarized, $\Delta R/R$ is a function of $\theta$ with a period of 180${}^{\circ }$. The data are fitted using the following equation:

$$\frac{\Delta R}{R}\left(\theta \right)=\frac{\Delta R_{\mathrm{iso}}}{R}+\frac{\Delta R_{\mathrm{ani}}}{R}\cos (2\theta -2{\theta }_0),$$

(1)

where $\Delta R_{\mathrm{ani}}/R$ and $\Delta R_{\mathrm{iso}}/R$ are anisotropic and isotropic transients, respectively, and ${\theta }_0$ is a phase corresponding to a direction wherein the transient signal is most enhanced. If the CO state appears, polarization dependence will change across the transition temperature. Even in that case, this analysis can characterize the anisotropy of the CO state as a change in ${\theta }_0$ [22]. Figure 3a,b show $\Delta R_{\mathrm{ani}}/R$ and $\Delta R_{\mathrm{iso}}/R$, respectively, for T = 20, 40, 80, 120, and 150 K. When the temperature decreases, the negative signal seems to increase in both components. We note that the double peak structure observed before ∼1.5 ps of the isotropic component is attributed to the oscillatory component. However, its origin is beyond the scope of this paper and is not discussed further.

To discuss the temperature dependencies in more detail, the data are fitted with a single exponential function

$$\frac{\Delta R_{\mathrm{ani}}}{R}\left(t\right)=A_{\mathrm{ani}}exp(-t{\tau }_{\mathrm{ani}})+C_{\mathrm{ani}}$$

(2)

for the anisotropic component or

$$\frac{\Delta R_{\mathrm{iso}}}{R}\left(t\right)=A_{\mathrm{iso}}exp(-t{\tau }_{\mathrm{iso}})+C_{\mathrm{iso}},$$

(3)

for the isotropic component, where $A_{\mathrm{ani}}$, $A_{\mathrm{iso}}$ and ${\tau }_{\mathrm{ani}}$, ${\tau }_{\mathrm{iso}}$ are the amplitude and relaxation time of a short-lived component. $C_{\mathrm{ani}}$ and $C_{\mathrm{iso}}$ are the amplitude of long-lived component when its relaxation time is assumed to be infinite. Figure 4a shows the temperature dependencies of the absolute values of $A_{\mathrm{ani}}$ and $C_{\mathrm{ani}}$. As temperature decreases, $|A_{\mathrm{ani}}|$ increases below $T^{\prime }$ = 50 K, which agrees with $T_{\mathrm{MI}}$. On the other hand, the temperature dependence of $|C_{\mathrm{ani}}|$ shows little change. Moreover, the ${\tau }_{\mathrm{ani}}$ values gradually reach ∼1.5 ps at low temperatures and show no significant change around $T^{\prime }$, as shown in Figure 4b. Figure 4c shows the temperature dependence of ${\theta }_0$ at a delay of 1 ps. The ${\theta }_0$ values are ∼135${}^{\circ }$ in the whole temperature range, indicating no anisotropic electronic ordering below $T^{\prime }$.

In the isotropic component, the temperature dependencies of $|A_{\mathrm{iso}}|$ and ${\tau }_{\mathrm{iso}}$ are similar to those in the anisotropic component. The similarity between the anisotropic and isotropic dynamics suggests that they have the same origin. We note a broad peak structure in the temperature dependencies of $A_{\mathrm{ani}}$ and $A_{\mathrm{iso}}$ at high temperatures, as shown in Figure 4a,d. This is due to a change in beam irradiation position with temperature variation and is not intrinsic.

Since the observed changes in $|A_{\mathrm{ani}}|$ and $|A_{\mathrm{iso}}|$ reflect the changes in non-equilibrium carrier distribution, information on the gap magnitude can be extracted from the temperature dependencies of $|A_{\mathrm{ani}}|$ and $|A_{\mathrm{iso}}|$. The gap (${\Delta }_{\mathrm{gap}}$) can be estimated by fitting with a temperature-independent gap model, which is often used in the gradual temperature dependence in the amplitude (A) such as pseudogap response in cuprate superconductors [25]. In the model, the amplitude is written as

$$A\left(T\right)\propto {\left[1+bexp\left(-\frac{{\Delta }_{\mathrm{gap}}}{k_{B}T}\right)\right]}^{-1},$$

(4)

where b, and $k_B$ are variable parameters for the fit and the Boltzmann constant, respectively. As shown by the dashed lines in Figure 4a,d, the data are fitted well, and the gap is estimated as ${\Delta }_{\mathrm{gap}}$≈ 24 meV and 35 meV for the anisotropic and the isotropic components, respectively, which agree with that estimated from the analysis of the Arrhenius plot in the resistivity measurements. Therefore, the results indicate that a band gap opens at $T^{\prime }$ = 50 K in the $\alpha$-BETS.

4. Discussion

Here, possible origins of the observed dynamics below $T^{\prime }$ are discussed through comparison with the isostructural salt $\alpha$-ET, which undergoes a CO transition at $T_{\mathrm{co}}$ = 135 K [26,27,28,29,30]. The CO state is characterized by three features of photoinduced carrier dynamics [22]. The first one is the signal amplitude, which begins to change at around $T_{\mathrm{co}}$, and the change is explained by the insulating gap formation due to the CO. Secondly, a divergent behavior of the relaxation time is observed just below $T_{\mathrm{co}}$. This behavior is attributed to a phonon-bottleneck effect [25] due to critical fluctuation related to long-range electronic ordering just below $T_{\mathrm{co}}$. Thirdly, ${\theta }_0$ changes to 90${}^{\circ }$ where the transient signal is most enhanced along the $\frac{1}{2}$(a + b) axis, below $T_{\mathrm{co}}$. This polarization anisotropy indicates an anisotropic ordering of electrons [31,32,33], consistent with the CO state.

In $\alpha$-BETS, the signal amplitude increases below $T^{\prime }$ = 50 K, which is similar to $\alpha$-ET. Considering the consistency between the pump–probe and resistivity measurements, this behavior can be attributed to the formation of an insulating gap. However, in contrast to $\alpha$-ET, there are no significant changes in ${\tau }_{\mathrm{ani}}$, ${\tau }_{\mathrm{iso}}$ and ${\theta }_0$ at $T^{\prime }$. The difference between $\alpha$-BETS and $\alpha$-ET suggests that the origin of the resistivity increase below $T^{\prime }$ differs from the CO state.

One of the possible origins of this is topological insulators (TIs), which generally have an insulator-type band gap in the bulk but have a gapless conducting phase on their surface. As shown in Figure 1a, the BETS molecule is obtained by replacing four inner sulfur atoms of the ET molecule with selenium atoms. Due to the fact that a spin-orbit coupling (SOC) increases with the selenium substitution, the SOC in $\alpha$-BETS can be more significant than in $\alpha$-ET. Indeed, a recent theoretical study has suggested that SOC induces a gap, leading to a weak topological insulator [7]. Moreover, electron correlation is also crucial for the emergence of the topological phase [12,13], and anomalous transport properties originating from correlation-induced topological insulators have been observed experimentally [19]. We comment on the difficulty to refer to the relation between the electron correlation anisotropy and the polarization anisotropy in $\Delta R/R$. The previous study indicated that the charge gap formation is due to the development of one-dimensional anisotropy of spin correlations [13]. However, it is difficult to refer to the relation because the polarization anisotropy in $\Delta R/R$ is a consequence of the anisotropy regarding the optical transitions after the pump irradiation and is not directly related to the low-energy electronic gap structure [21].

In TI states, there is no anisotropy due to charge disproportionation. This means that the dynamics of the state are expected to stay constant with the relaxation time and ${\theta }_0$, and only the amplitude is likely to vary due to the bulk gap. These predictions are consistent with the present results, suggesting that the dynamics observed below $T^{\prime }$ = 50 K could be due to the insulator gap as a bulk property of TI. It is also worth noting that the present results do not show any anomaly in dynamics at around 40 K, where the resistivity shows a step-like change [11]. The recent study has suggested a crossover from two-dimensional to three-dimensional TI at ∼35 K [19], resulting in a change in the conducting surface states. Therefore, during the crossover, the bulk band gap is not affected, which is consistent with the lack of change in dynamics. In general, it is difficult to distinguish between the carrier dynamics arising from the bulk state and those from the surface state. Thus, other measurements, such as a spectrally resolved pump–probe measurements, may be needed to clarify the contribution from the surface.

5. Conclusions

Through pump–probe time-resolved spectroscopy, the photo-induced carrier dynamics were found to change below $T^{\prime }$ = 50 K. This finding corresponds to the increase in resistivity. Compared with $\alpha$-ET, the observed dynamics below $T^{\prime }$ differ from those in the CO state regarding relaxation time and polarization anisotropy, but they are compatible with those predicted in the TI.