Negative terahertz conductivity in disordered graphene bilayers with population inversion

Negative terahertz conductivity in disordered graphene bilayers with population inversion

Abstract

The gapless energy band spectra make the structures based on graphene and graphene bilayers with the population inversion created by optical or injection pumping to be promising media for the interband terahertz (THz) lasing. However, a strong intraband absorption at THz frequencies still poses a challenge for efficient THz lasing. In this paper, we show that in the pumped graphene bilayer structures, the indirect interband radiative transitions accompanied by scattering of carriers caused by disorder can provide a substantial negative contribution to the THz conductivity (together with the direct interband transitions). In the graphene bilayer structures on high- substrates with point charged defects, these transitions almost fully compensate the losses due to the intraband (Drude) absorption. We also demonstrate that the indirect interband contribution to the THz conductivity in a graphene bilayer with the extended defects (such as the charged impurity clusters, surface corrugation, and nanoholes) can surpass by several times the fundamental limit associated with the direct interband transitions and the Drude conductivity. These predictions can affect the strategy of the graphene-based THz laser implementation.

The absence of a band gap in the atomically thin carbon structures,such as graphene and graphene bilayers, enables their applications in different terahertz (THz) and infrared devices (1); (2); (3); (4). One of the most challenging and promising problems is the creation of the graphene-based THz lasers (5); (6); (7). These lasers are expected to operate at room temperature, particularly, in the 6-10 THz range, where the operation of III-V quantum cascade lasers is hindered by the optical phonons (8). Recent pump-probe spectroscopy experiments confirm the possibility of the coherent radiation amplification in the optically pumped graphene (9); (10); (11); (12); (13); (14); (15); (16), enabled by a relatively long-living interband population inversion (17). As opposed to optically pumped graphene lasers, graphene-based injection lasers are expected to operate in the continuous mode, with the interband population inversion maintained by the electron and hole injection from the - and -type contacts (18). A single pumped graphene sheet as the gain medium provides the maximum radiation amplification coefficient corresponding to the quantity , where is the universal optical conductivity of a single graphene layer, is the electron charge, is the Planck constant and is the fine-structure constant (17). The THz gain in the graphene bilayers (19) or the non-Bernal stacked multiple-graphene layers (5) can be enhanced approximately proportional to the number of the layers. However, more crucial is the problem of competition between the interband radiation amplfication and intraband (Drude) radiation absorption (17); (20). The latter scales with frequency approximately as , where is the momentum relaxation time. Hence, the onset of terahertz gain is typically believed to occur only in clean samples, where  (21).

Figure 1: Energy band diagram of a graphene bilayer with population inversion (left) and schematic energy dependence of its density of states (right). Direct interband transitions involve only vertical photon emission (wavy arrow), while indirect emission and absorption processes are accompanied by carrier scattering (straight horizontal arrows).

In this letter, we show that the intraband radiation absorption in disordered graphene bilayers does not actually pose a problem for the THz lasing. On the contrary, the presence of a certain type of defects reinforces the negative contribution to the THz conductivity and, hence, improves the gain properties of the pumped graphene bilayers. The origin of such an effect is associated with the indirect interband radiative transitions (see Fig. 1), in which the electrons from the conduction band emit the photons being scattered on the defects, thus contributing to the radiation gain. The inclusion of such processes can be important in the indirect-gap materials and gapless semiconductors. However, in single-layer graphene with charged impurities, the indirect interband processes contribute to the net THz conductivity only moderately due to a low density of states (DoS) near the band edges (except, possibly, for the case of the carrier interactions with artificial fairly large-size scatterers (22)) . The situation is remarkably different is the intrinsic graphene bilayers, where the electron-hole dispersion is gapless and almost parabolic (23). With constant DoS near the band edges, the indirect interband radiative processes significantly contribute to the net radiation gain under the population inversion conditions. The THz gain is proportional to . We analyze the spectral dependencies of the real part of the net dynamic THz conductivity in the pumped graphene bilayers for the scattering by the point charged impurities (24); (25) and by the impurity clusters (26); (27). Our analysis shows that in the first case, the gain due to the indirect interband transition almost fully compensates the losses due to the Drude absorption. In the case of the cluster scattering, the gain he indirect interband transitions exceeds the intraband losses. Depending on the cluster size and their density, the ratio can markedly exceed unity resulting elevated net THz gain.

The real part of the net in-plane dynamic THz conductivity, , comprises the contributions of the direct (vertical) interband electron transitions, , and the contributions, and , of two types of the indirect electron transitions (inside both the bands and between the two bands), respectively:

(1)

The interband conductivity of graphene bilayers due to the direct transitions is given by (19); (23)

(2)

where and are the carrier distribution functions in the valence and conduction bands, and  eV is the hopping integral between carbon atoms in adjacent graphene planes (28). Here and in the following, for the intrisic graphene bilayers we assume and are the Fermi functions characterized by the quasi-Fermi energies and , respectively. This is justified by strong carrier-carrier scattering leading to a fast thermalization of excited carriers (9); (13). In the THz frequency range of interest, , and the conductivivty of bilayer is simply twice as large as that for a single layer. Under the pumping conditions, , and, according to Eq. (2), the THz conductivity is negative for photon energies below the double quasi-Fermi energy of pumped carriers (17).

To evaluate the real part of the THz conductivity due to the indirect transitions, we calculate the second-order transition amplitudes for the photon emission (absorption) accompanied by the electron scattering and apply the Fermi’s golden rule. As a result, the general expressions for the indirect intra- and interband THz conductivities read as follows:

(3)
(4)

Here is the index corresponding to the conduction and valence bands, is the electron velocity in the graphene bilayer, cm/s is the velocity characterizing the energy spectra of graphene and graphene bilayers. is the -th Fourier component of the scattering potential, and is the overlap between the envelope wave functions in graphene bilayers. Equation (3) reproduces the well-known result for the dynamic conductivity in the high-frequency limit , where is the momentum relaxation time, which can be derived from the Boltzmann equation. For a correct qualitative description of the low-frequency conductivity, we replace the frequency in the denominators of Eqs. (2) and (3) with .

In the most practical situations,the Coulomb scattering by the random substrate-induced charged impurities is the main factor determining the conductivity (29). Considering impurities as random uncorrelated point scatterers with the average density , we write the scattering matrix element as (30)

(5)

where is the background dielectric constant, and is the Thomas-Fermi screening wave vector (30). In the case of the interband population inversion, the latter is found to be , where is the coupling constant. Evaluating the integral, we find the scattering-assisted interband conductivity

Figure 2: Contributions of different radiative transitions to dynamic THz conductivity of a graphene bilayer on SiO () and its net value (solid line) versus frequency for cm and meV (upper panel), and color map (bottom panel). Numbers above the lines indicate the values of . The region above dashed line corresponds to the negative conductivity.
Figure 3: The same as in Fig. 2 but for graphene bilayer clad by Hf0 layers ().
(6)

where with the following asymptotes: , , , . At intermediate frequencies, , the conductivity due to the indirect interband transitions scales as . This is substantially different from the case of a single graphene layer, where it tends to a constant. A pronounced increase in the indirect interband contribution to the dynamic conductivity in a bilayer at low frequencies is attributed to the constant density of states in the vicinity of the band edges.

Figure 2 (upper panel) shows the spectral dependencies of the contributions of different radiative transitions to the dynamic THz conductivity as well the net value of the latter for a moderate-quality exfoliated graphene bilayer  (25) on the SiO substrate with the effective dielectric constant (graphene bilayer sandwiched between SiO and air) impurity density  cm, at temperature  K, and for the quasi-Fermi energy  meV. The bottom panel in Fig. 2 demonstrates the two-dimensional maps of the dynamic THz conductivity versus the frequency and the quasi-Fermi energy for the same structure. As seen, the contribution of the indirect interband transitions in such a sample is weaker than those of both the indirect intraband and direct interband transitions, although the former is essential for compensating, to some extend, the Drude absorption. This enables an increase in and some widening of the frequency range where . As follows from Fig. 2 (bottom panel), the dynamic THz conductivity is negative at  meV and  THz.

The relative contribution of the indirect interband transitions(compared to the ”normal” intraband conductivity) increases with an increasing dielectric constant. Figure 3 shows the same characteristics as in Fig. 2, for a graphene bilayer being clad by the HfO layers, i.e., immersed in a media with a fairly high dielectric constant (). As seen from Fig. 3, the transition to the graphene bilayer structures with higher dielectric constant leads to a much stronger contribution of the indirect interband transitions and, hence, to a much larger value of . The comparison of Figs. 2 and 3 shows that the ratio for the minimum value of of at is five-six time larger than for . Moreover, in the former case becomes negative starting from  meV and  THz. At higher values of (i.e., at a stronger pumping), can be negative from the frequencies of about a few THz to a dozen THz.

The reinforcement of the negative dynamic THz conductivity effect with increasing background dielectric constant demonstrated above is interpreted as follows. An increase in results in the reduced Thomas-Fermi wave vector . This, in turn, leads to switching from the strongly screened to almost bare Coulomb scattering. From the energy conservation laws it follows that the indirect interband electron transitions are favored by a low momentum transfer , while for the indirect transitions within one band should be large, namely, as the electron velocity in GBL does not exceed . Hence, for high values of , the scattering potential behaves approximately as , which supports the interband transitions with a low momentum transfer.

Figure 4: Net THz conductivity vesus frequency calculated for graphene bilayers on SiO with impurity clusters of different size : cluster density and charge are  cm and , dielectric constant , and quasi-Fermi energy  meV. Dashed line corresponds to point charged defects with the same charge and density.

As shown above, the Coulomb scattering by the screened point defects cannot lead to the dominance of the indirect interband transitions over the indirect intraband ones. However, such a dominance can be realized in the case of the carrier scattering on sufficiently extended scatterers. We consider the charged cluster of size and charge as a continuous two-dimensional distribution of charge density (since the exact density distribution is not very important, for simplicity, we assume it to be Gaussian (27)). Solving the Poisson equation for this charge density and averaging over the random positions of the clusters, we readily find the scattering matrix elements [instead of Eq. (5)]

(7)

Here is the density of the clusters. In the limit of strong screening, , our model of scattering coincides with the widely accepted model of the ”Gaussian correlated disorder” (31); (32); (33); (34) with the root-mean-square scattering potential .

Figure 4 shows the spectral characteristics of the dynamic THz conductivity in the pumped graphene bilayers ( meV) with clusters of charged impurities with different size . If the scattering by the charged clusters is a dominating mechanism, the absolute value of the net dynamic THz conductivity can markedly exceed the fundamental ”direct interband limit” of . At reasonable values of nm and quasi-Fermi energy meV, one obtains .

In conclusion, we have demonstrated that the graphene bilayers with a long-range disorder (impurity clusters with reasonable values of the cluster density and size), can exhibit a strong negative THz conductivity with the span two times or more exceeding the fundamental limit . This effect is associated with the indirect interband transitions with the photon emission being accompanied by the disorder scattering. For the indirect interband photon emission to dominate over the ”normal” Drude absorption, the long-wave length Fourier components of the scattering potential should prevail. Such kind of scattering potentials can be formed also by extended surface corrugations, quantum dots on the graphene bilayer surface (35), and nanohole arrays (36); (37).

The work was supported by the Japan Society for Promotion of Science (Grant-in-Aid for Specially Promoted Research 23000008) and by the Russian Scientific Foundation (Project 14-29-00277) and the grant of the Russian Foundation of Basic Research 14-07-31315. The works at UP and RPI were supported by the US Air Force award FA9550-10-1-391 and by the US Army Research Laboratory Cooperative Research Agreement, respectively.

Footnotes

  1. Electronic mail: v-ryzhii(at)riec.tohoku.ac.jp

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