Independent Dual-Channel Approach to Mesoscopic Graphene Transistors

Abstract

Graphene field-effect transistors (GFETs) exhibit unique switch and sensing features. In this article, GFETs are investigated within the tight-binding formalism, including quantum capacitance correction, where the graphene ribbons with reconstructed armchair edges are mapped into a set of independent dual channels through a unitary transformation. A new transfer matrix method is further developed to analyze the electron transport in each dual channel under a back gate voltage, while the electronic density of states of graphene ribbons with transversal dislocations are calculated using the retarded Green’s function and a novel real-space renormalization method. The Landauer electrical conductance obtained from these transfer matrices was confirmed by the Kubo–Greenwood formula, and the numerical results for the limiting cases were verified on the basis of analytical results. Finally, the size- and gate-voltage-dependent source-drain currents in GFETs are calculated, whose results are compared with the experimental data.

1. Introduction

Graphene is a one-atom-thick planar sheet of carbon atoms in a honeycomb structure, whose free-standing monolayer was isolated and characterized for the first time in 2004 by Andre Geim and Konstantin Novoselov [1]. This material possesses outstanding properties such as high specific surface area [2], very high carrier mobility with null effective mass [3], huge thermal conductivity, and giant Young’s modulus [4], making it an ideal candidate for a wide range of applications [5].

When the semiconductor layer of a traditional metal–oxide–semiconductor field-effect transistor (MOSFET) is replaced by a graphene sheet, it is called as graphene field-effect transistor (GFET), whose source-drain current is extremely sensitive to the adsorbed molecules, and it is employable for use in gas and bio sensing [6,7,8]. Moreover, GFET constitutes a central component of far-infrared radiation and terahertz devices [9] since graphene exhibits a quick optical response based on high carrier mobility [10]. In addition, the graphene nanoribbon field-effect transistor (GNRFET) presents an elevated $I_{on}/I_{off}$ ratio around the threshold voltage compared to the conventional Si-based CMOS [11]. Among possible disadvantages of GFETs, there are difficulties in fabricating wafer-sized high-quality graphene, as well as the apparent degradation of carrier mobility when it is placed over an oxide [12].

Additionally, GFET has a singular capacitor behavior, since the graphene ribbon, being one of the parallel plates, possesses a very low charge density around the Dirac point, which may induce large variations in its chemical potential when a small amount of electric charge is introduced into the capacitor. This fact could significantly increase the potential difference between the back gate and the graphene, because it is equal to the difference between the chemical potentials at each plate. Such small quantities of charge generating a large potential difference lead to a lower capacitance compared to geometric or classic ones ($C_C$) obtained using ideal metal plates. Hence, the capacitance of GFET $(C_{tot})$ can be calculated by including a so-called quantum capacitance ($C_Q$) through $C_{tot}^{-1}=C_C^{-1}+C_Q^{-1}$ [13].

On the theoretical side, GFETs can be modeled at the atomic scale by means of first-principle or semiempirical methods. For example, N/B/P co-doped seven-atom-wide armchair GNRFET was analyzed by using the density functional theory (DFT) [14], while ten-atom-width GNRFET has been studied by self-consistently solving Schrödinger–Poison equations within the tight-binding formalism [15]. Recently, mesoscopic GFETs have been extensively investigated for the detection of micron-scale biomolecules [16] and their graphene ribbons contain several billions of atoms, which impede atomic-scale first-principle modeling. In addition, such graphene ribbons usually possess numerous structural defects, which requires an innovative real-space approach [17].

In this article, the source-drain current ($I_{sd}$) in mesoscopic GFETs is studied by means of an independent dual-channel method that transforms the graphene ribbon with edge reconstruction defects and transversal dislocations into a set of double chains with first and second neighbor interactions within the tight-binding formalism. The electrical conductance and electronic density of states in these double chains or dual channels connected to two semi-infinite periodic leads at their ends are further addressed by means of a new transfer matrix method within the Landauer formalism and a novel real-space renormalization procedure based on the retarded Green’s function, respectively. The theoretical $I_{sd}$, as a function of the gate voltage, is compared with experimental data obtained from GFETs of different lengths.

2. The Model

In GFETs, an extra carrier density ($n_{2D}$) can be induced in graphene ribbon by the application of a gate voltage ($V_G$), which is related to the chemical potentials of graphene ($\mu$) and of back gate metal (${\mu }_M$) through $e{V}_G=\mu -{\mu }_M$. Figure 1 shows a schematic representation of (Figure 1a) top and (Figure 1b,c) side views of a backgated GFET with energy band diagrams for (b) $V_G=0$ and (c) $V_G>0$, where the diminution of ${\mu }_M$ due to $V_G$ is denoted as $e{V}_C$. Hence, we have:

$$e{V}_G=\mu -{\mu }_M=\mu +e{V}_C,$$

(1)

which is equivalent to $C_{tot}^{-1}=C_C^{-1}+C_Q^{-1}$, since $C_{tot}=e \partial n/\partial V_G$, $C_C=e \partial n/\partial V_C$, $C_Q=e \partial n/\partial V_Q$ and $e V_Q=\mu -{\mu }_0$ with ${\mu }_0=0$ or at the Dirac point in our case [18].

In general, the capacitance per unit of area (C) of an ideal parallel-plate capacitor with a dielectric material of thickness d and a relative permittivity ${\epsilon }_r$ is $C={\epsilon }_r{\epsilon }_0/d=Q/V_C$ in units of MKS [19], where ${\epsilon }_0$ is the vacuum permittivity, $Q=e{n}_{2D}$ is the electric charge per unit of area in the capacitor and $V_C$ is the potential difference between the parallel plates. Hence:

$$e{V}_C=\frac{e^2{n}_{2D}d}{{\epsilon }_r{\epsilon }_0},$$

(2)

where e is the magnitude of the electron charge.

Let us consider an armchair-edged graphene ribbon with an even number of atoms (2W) in each transversal zig-zag line, as illustrated in Figure 2a. This ribbon of width $\mathcal{W} =\sqrt{3}{a}_S+\sqrt{3}(2W-3) a_0/2$ and length $\mathcal{L}=(3/2)L{a}_0-a_0$ is found in a backgated GFET, where W and L are integer numbers, $a_0=1.41$ Å and $a_S=1.36$ Å are bond lengths between interior atoms and between the edge and next-edge atoms, respectively denoted by blue and thick blue lines in Figure 2a. This variation in interatomic distance is originated from the edge reconstruction of graphene ribbons [20]. The single-electron tight-binding Hamiltonian (H) of this graphene ribbon with null on-site energies can be written as

$$\begin{array}{cc}H=\hfill & \hfill {\displaystyle \sum _{l = 1}^L\left(t_s\left|l,1\right.〉\left.〈l,2\right|+t{\displaystyle \sum _{j = 2}^{2W-2}\left|l,j\right.〉\left.〈l,j+1\right|}+t_s\left|l,2W-1\right.〉\left.〈l,2W\right|\right)}\\ \hspace{1em}+\hfill & \hfill {\displaystyle \sum _{l = 1}^{(L-1)/2}{\displaystyle \sum _{j = 1}^W\left(t_{2l-1}\left|2l-1,2j\right.〉\left.〈2l,2j\right|+t_{2l}\left|2l,2j-1\right.〉\left.〈2l+1,2j-1\right|\right)}},\end{array}$$

(3)

where $\left|l,j\right.〉$ is the Wannier function at site $(l,j)$, t is the hopping integral of pristine graphene sheet and $t_s =1.2 t$ is that between the edge and next-edge atoms in a graphene ribbon with edge reconstructions [20] and $t_l$ with $l=1,\hspace{0.33em}2,\hspace{0.33em}\cdots ,\hspace{0.33em}L-1$ is the hopping integral between transversal zig-zag lines l and $l+1$, representing possible transversal dislocations when $t_l \ne t$.

There is a unitary transformation discussed in Appendix A that converts the Hamiltonian (3), including the edge reconstruction defects, into a set of W independent dual channels, whose Hamiltonian contains hopping integrals $t^{\prime } =t/2$, ${t^{\prime }}_l =t_l/2$ with $l=1,\hspace{0.33em}2,\hspace{0.33em}\cdots ,\hspace{0.33em}L-1$ and on-site energies $\pm {\epsilon }_j$ with $j=1, 2,\cdots , W,$ which are eigenvalues obtained from the Hamiltonian of an arbitrary transversal zig-zag line in Figure 2.

The extra carrier density ($n_{2D}$) induced by $V_G$ in the graphene ribbon can be calculated by [21]

$$n_{2D}={\displaystyle {\int }_{ 0}^{\mu }DOS(E)} dE={\displaystyle {\int }_0^{e{V}_G- e{V}_C}DOS(E)} dE,$$

(4)

where

$$DOS(E)=-\frac{1}{\pi }\mathrm{Im}\left\{Tr [G^{+}(E)]\right\},$$

(5)

is the density of states with $G^{+}(E) =\underset{\eta \hspace{0.33em}\to 0^{+}}{\lim }{(E+i\eta -H)}^{-1}$ the retarded Green’s function and η the imaginary part of energy [22]. Combining Equations (2) and (4), $V_C$ can be determined as the solution of following self-consistent equation,

$$e{V}_C =\frac{e^{2}d}{{\epsilon }_r{\epsilon }_0}{\displaystyle {\int }_0^{e{V}_G- e{V}_C}DOS(E)} dE.$$

(6)

On the other hand, the source-drain current ($I_{sd}$) of GFETs at temperature T is given by [23]

$$I_{sd}(T)=V_{sd}\mathrm{g}(\mu ,T),$$

(7)

where $V_{sd}$ is the source-drain voltage and

$$\mathrm{g}(\mu ,T)={\displaystyle {\int }_{-\infty }^{+\infty }dE\left(-\frac{\partial f_{FD}(E)}{\partial E}\right)}\hspace{0.33em}\mathrm{g}(E,0)={\mathrm{g}}_0{\displaystyle {\int }_{-\infty }^{+\infty }dE\left(-\frac{\partial f_{FD}(E)}{\partial E}\right)} \mathrm{T}(E)$$

(8)

is the electrical conductance of graphene ribbon at chemical potential μ within the Landauer formalism. In Equation (8), $f_{FD}={\{\exp [(E-\mu )/k_{B}T]+1\}}^{-1}$ is the Fermi–Dirac distribution, ${\mathrm{g}}_0=2e^2/h$ is the conductance quantum, $\mathrm{T}(E)$ is the carrier transmittance of graphene ribbon, and at zero temperature we have [24]

$$\mathrm{g}(\mu ,0)={\mathrm{g}}_0\mathrm{T}(\mu ).$$

(9)

By means of the independent dual-channel method presented in Appendix A, an armchair-edged graphene ribbon can be transformed into a set of double chains or dual channels (see Figure 2) and then

$$\mathrm{T}(E)={\displaystyle \sum _{j=1}^W{\mathrm{T}}_j(E)},$$

(10)

where ${\mathrm{T}}_j(E)$ is the carrier transmittance along the j-th dual channel. We further developed a new transfer matrix method to calculate ${\mathrm{T}}_j(E)$, which is thoroughly presented in Appendix B, and the result can be written as

$${\mathrm{T}}_j(E)={\left|\frac{u_0(j) d_0^{\ast }(j)-d_0(j) u_0^{\ast }(j)}{m_{11}(j,E) d_0(j) u_0^{\ast }(j)+m_{12}(j,E)|d_0(j) {|}^2- m_{21}(j,E) |u_0(j) {|}^2- m_{22}(j,E) u_0(j) d_0^{\ast }(j)}\right|}^2,$$

(11)

where $m_{\mu \nu }(j,E)$ are elements of the total transfer matrix, $u_0(j)$ and $d_0(j)$ are respectively initial wavefunction amplitudes at the up and down channels, both from the j-th dual channel (see Appendix B).

One of structural defects commonly observed in graphene ribbons is linear dislocation [25,26], because its presence slightly alters the free energy but may significantly modify the carrier transport. In this article, we consider a distribution of transversal dislocations following the Rudin–Shapiro (RS) sequence, which constitutes one of the closest aperiodic arrays to the random distribution [27]. A Rudin–Shapiro lattice with bond disorder can be built by using four kinds of dislocation hopping integrals $t_l=t_A, t_B, t_C \mathrm{or} t_D$, respectively denoted by letters A, B, C or D, whose positions along the ribbon are ordered by the substitution rules [28]

$$A\to A\oplus B=AB,\hspace{1em}B\to A\oplus C=AC,\hspace{1em}C\to D\oplus B=DB,\hspace{1em}D\to D\oplus C=DC$$

(12)

or by the addition rules expressed as

$$\begin{array}{l}{S}_A(k+1)=S_A(k)\oplus S_B(k), S_B(k+1)=S_A(k)\oplus S_C(k), \\ S_C(k+1)= S_D(k)\oplus S_B(k), S_D(k+1)= S_D(k)\oplus S_C(k),\end{array}$$

(13)

where the symbol $\oplus$ represents the concatenation operation and $S_{\alpha }(k)$ is the α-type RS sequence of generation k with $\alpha = A,B,C \mathrm{or} D$. As a consequence, a graphene ribbon based on $S_{\alpha }(k)$ has $2^k+1$ transversal zig-zag lines. To have a limited number of dislocations, let us introduce dilute RS lattices, which are built by using periodic segments to construct the RS lattice until generation $m-1$ and a single transversal dislocation is placed at the initial of next generation m. For example, when $k=m=3$, $S_A(3)=APPP$, $S_B(3)=BPPP$, $S_C(3)=CPPP$ and $S_D(3)=DPPP$, where P denotes a periodic RS sequence with hopping integral t connecting all transversal zig-zag lines. A detailed discussion of this dilute RS lattice and the real-space renormalization method can be found in Appendix C.

Another quantity that should be considered for determining the electrical conductance is the contact resistance between the graphene ribbon and periodic leads. In the diffusive regime, the total resistance ($R_{total}$) can be written as [29,30]

$$R_{total}=R+2R_c/\mathcal{W},$$

(14)

where $R=R_{sheet}\mathcal{L}/\mathcal{W}$ is the electrical resistance of a graphene ribbon with length $\mathcal{L}$ and width $\mathcal{W}$, being $R_{sheet}$ that of a square graphene sheet, and $R_c$ is the specific contact resistance in units of $\Omega ·$ μm, which can be experimentally determined by the transfer length method [31]. Hence, the total conductance defined as $G_{total}=R_{total}^{-1}$ can be calculated from Equation (14) through

$$G_{total}=\frac{G}{2(R_c/\mathcal{W}) G+1},$$

(15)

where $G=R^{-1}$ is the conductance of graphene ribbon. For a uniform sample, the electrical resistance of a p-micron segment, R($\mathcal{L}=p$ μm), should be $p/q$ times of R($\mathcal{L}=q$ μm) obtained from a q micrometer portion. Therefore, Equation (15) can be rewritten as

$$G_{total}(p \mathsf{\mu }\mathrm{m})=\frac{G(p \mathsf{\mu }\mathrm{m})}{2(R_c/\mathcal{W}) G(p \mathsf{\mu }\mathrm{m})+1}=\frac{G(q \mathsf{\mu }\mathrm{m})}{2(R_c/\mathcal{W}) G(q \mathsf{\mu }\mathrm{m})+p/q},$$

(16)

where $G(p\hspace{0.33em}\mathsf{\mu }\mathrm{m})=qG(q\hspace{0.33em}\mathsf{\mu }\mathrm{m})/p$. This equation will be used in the length variation analysis.

3. Results

The electronic density of states, $DO{S}^{\alpha }(k,E)$, of a graphene ribbon built by W dual channels based on an α-type dilute RS sequence of generation k can be written as [22]

$$DO{S}^{\alpha }(k,E)={\displaystyle \sum _{j=1}^{W}DO{S}_j^{\alpha }(k,E)}={\displaystyle \sum _{j=1}^W\left\{-\frac{1}{\pi }\underset{\eta \hspace{0.33em}\to \hspace{0.33em}{0}^{+}}{\lim }{\displaystyle \sum _{l=1}^{L(k)}\mathrm{Im} [G_{l,l}^{\alpha ,j}(k,z)}]\right\}},$$

(17)

where $L(k)=2 (2^k+1)$ is the number of sites in each dual channel and $G_{l,l}^{\alpha ,j}(k,z)$ is the l-th diagonal element of the retarded Green’s function evaluated at $z=E+i\eta$. The $DO{S}_j^{\alpha }(k,E)$ of the j-th dual channel can be rewritten as

$$\begin{array}{c}DO{S}_j^{\alpha }(k,E)=-\frac{1}{\pi }\underset{\eta \hspace{0.33em}\to \hspace{0.33em}{0}^{+}}{\lim }\mathrm{Im} \left[M^{\alpha }(k) G_{L,L}^{\alpha ,j}(k,z) +P^{\alpha }(k) G_{\underset{\_}{L},\underset{\_}{L}}^{\alpha ,j}(k,z) + Q^{\alpha }(k) G_{R,R}^{\alpha ,j}(k,z) \right.\hfill \\ \hspace{1em}\hspace{1em}\hspace{1em}\hspace{1em}\hspace{1em}+ R^{\alpha }(k) G_{\underset{\_}{R},\underset{\_}{R}}^{\alpha ,j}(k,z) +S^{\alpha }(k) G_{L,\underset{\_}{L}}^{\alpha ,j}(k,z)+U^{\alpha }(k) G_{L,R}^{\alpha ,j}(k,z)+V^{\alpha }(k) G_{L,\underset{\_}{R}}^{\alpha ,j}(k,z)\hfill \\ \hspace{1em}\hspace{1em}\hspace{1em}\hspace{1em}\hspace{1em}\left.+\hspace{0.33em}{W}^{\alpha }(k) G_{\underset{\_}{L},R}^{\alpha ,j}(k,z)+ X^{\alpha }(k) G_{\underset{\_}{L},\underset{\_}{R}}^{\alpha ,j}(k,z)+Y^{\alpha }(k) G_{R,\underset{\_}{R}}^{\alpha ,j}(k,z)+Z^{\alpha }(k)\right],\hfill \end{array}$$

(18)

where $M^{\alpha }(k) ,\hspace{0.33em}\cdots \hspace{0.33em},\hspace{0.33em}{Z}^{\alpha }(k)$ are the renormalization coefficients and $G_{\mu ,\nu }^{\alpha ,j}(k,z)$ with $\mu ,\nu =L,\hspace{0.33em}\underset{\_}{L},\hspace{0.33em}R \mathrm{or} \underset{\_}{R}$ are matrix elements of the Green’s function corresponding to the left up (L), left down (L), right up (R) and right down (R) sites of the renormalized four-site j-th dual channel, which constitutes the basic element of the real-space renormalization method presented in Appendix C.

Figure 3 shows the electronic density of states (DOS) and the electrical conductance (g) at zero temperature in units of the conductance quantum ${\mathrm{g}}_0=2e^2/h$ obtained from Equation (9) as functions of the chemical potential (μ) for free-standing graphene ribbons without dislocations, whose widths are $\mathcal{W}=0.122 \mathsf{\mu }\mathrm{m}$ (red lines), $0.073 \mathsf{\mu }\mathrm{m}$ (dark yellow lines) and $0.037 \mathsf{\mu }\mathrm{m}$ (blue lines) as well as an arbitrary length of L transversal zig-zag lines. All the ribbons studied in this article are connected to two semi-infinite periodic leads at their ends, as illustrated in Figure 2a, while a surface hopping integral $t_s=1.2 t$ due to the edge reconstruction and an imaginary part of energy $\eta ={10}^{-3}| t |$ are also included.

Observe the Van Hove singularities in the inset of Figure 3a, which are located at the band limits of each dual channel. The DOS spectra of Figure 3a can be analytically verified through [32]

$$DOS(E)=\frac{dS/dk}{|dE/dk |}={\displaystyle \sum _{j= 1}^W\frac{2\left|E\right|}{\pi \sqrt{4t^2{\epsilon }_j^2-{(E^2-4t^2-{\epsilon }_j^2)}^2}}},$$

(19)

where $dS/dk=La/(2\pi )$ and $dE/dk$ can be obtained from Equation (A9) in Appendix B. Note also the quantized conductance spectra in the inset of Figure 3b and the maximum values of $\mathrm{g}(E,0)$ around $E=\pm t$ in Figure 3b is equal to the number of dual channels (W).

To analyze the electrical conductance (g) of GFETs, we first self-consistently calculate $V_C$ from Equation (6) for a given $V_G$ and then, the chemical potential μ and $\mathrm{g}$ can be respectively determined using Equations (1) and (8). Figure 4 shows the electrical conductance (g) at $T =0$ (blue lines) and at $k_{B}T=0.02| t |$ (red lines) versus the gate voltage ($V_G$) for GFETs of $\mathcal{W}=0.122 \mathsf{\mu }\mathrm{m}$, i.e., $W=500$ dual channels, and $L=4097$ zig-zag lines without dislocations, whose capacitances per unit area are (a) $C=10\hspace{0.33em}\mathrm{nF}/{\mathrm{cm}}^2$ and (b) $C=50\hspace{0.33em}\mathrm{nF}/{\mathrm{cm}}^2$. Note the quantized conductance spectra for $T =0$, in contrast to the smoothed ones when T increases, as well as the growth of conductance with the capacitance.

In Figure 5, the electrical conductance ($\mathrm{g}$) at $k_{B}T =0.026| t |$ is plotted as a function of both the back gate voltage $(V_G)$ and the dislocation hopping integral $t_A$ for the same graphene ribbon of Figure 4 except by the value of $t_A$ maintaining $t_B=t_C=t_D=t$. This ribbon contains 72 A-type transversal dislocation lines obtained from a A-type dilute RS lattice with $k=12$ and dislocations introduced from generation $m=5$, and it is placed on a GFET with a capacitance per unit area $C=10 \mathrm{nF}/{\mathrm{cm}}^2$. Observe the V-shaped dependence between g and $V_G$, even for $t_A=0.9 t$, and this dependence can be noted from Figure 3b, since $V_G$ modifies the value of chemical potential μ, as shown in Figure 1c.

Figure 6 shows the electrical conductance (g) at (Figure 6a) $k_{B}T=0.01\left|t\right|$ and (Figure 6b) $k_{B}T=0.02\left|t\right|$ with $t=-2.70 \mathrm{eV}$ [20] as functions of the gate voltage ($V_G$) for GFETs of $\mathcal{W}=0.122 \mathsf{\mu }\mathrm{m}$ (i.e., $W=500$ dual channels) and $\mathcal{L}=0.217 \mathsf{\mu }\mathrm{m}$ (red lines), $0.433 \mathsf{\mu }\mathrm{m}$ (green lines), and $0.866 \mathsf{\mu }\mathrm{m}$ (blue lines), respectively corresponding to generations $k=10$, 11 and 12 of A-type dilute RS sequences with dislocations introduced from generation $m=3$, hopping integrals $t_A=-2.389 \mathrm{eV}$, $t_B=t_C=-2.74 \mathrm{eV}$ and $t_D=-2.63 \mathrm{eV}$, where the capacitance per unit area of GFET is $C=10\hspace{0.33em}\mathrm{nF}/{\mathrm{cm}}^2$.

The results reveal a more emphasized V-shaped conductance behavior at lower temperatures, while the electrical conductance diminishes with increasing RS generation, being almost inversely proportional to the GFET length, in accordance with the Ohm’s law as well as the length variation measurements carried out in GFET [33].

Finally, let us consider a specific GFET [29] built by an armchair-edged graphene ribbon placed on a substrate of silicon dioxide (SiO₂) of thickness $d=285\hspace{0.33em}\mathrm{nm}$, i.e., a geometric capacitance per unit area of $C={\epsilon }_0{\epsilon }_r/d\approx 12.11\hspace{0.33em}\mathrm{nF}/{\mathrm{cm}}^2$. We first calculated the electrical conductance g of a graphene ribbon having a width of $W =9009$ dual channels ($\mathcal{W}=2.2 \mathsf{\mu }\mathrm{m}$) and a length of $L=4097$ zig-zag lines ($\mathcal{L}=0.866 \mathsf{\mu }\mathrm{m}$ corresponding to generation 12 of the RS sequence), which contains 1024 transversal dislocation lines from a A-type dilute RS lattice with $m=3$ and hopping integrals $t=-2.7 \mathrm{eV}$, $t_s=1.2 t$, $t_A=-2.389 \mathrm{eV}$, $t_B=t_C=-2.74 \mathrm{eV}$ and $t_D=-2.63 \mathrm{eV}$ as in Figure 6, while the analysis of system length ($\mathcal{L}$) effects on the conductance was carried out by means of Equation (16). Additionally, the contact resistance described in ref. [29] is included in the total conductance $(G_{total})$ using Equation (15). In Figure 7, we present the source-drain current ($I_{sd}$) at $T=300 \mathrm{K}$ as a function of the gate voltage $(V_G)$ and graphene ribbon length ($\mathcal{L}$) for the considered GFET with a source-drain voltage of $V_{sd} =0.05 \mathrm{volts}$, where $I_{sd}(T)$ (red spheres) was obtained from $I_{sd}=V_{sd}{G}_{total}$ and Equation (16) with $q=0.866\hspace{0.33em}\mathsf{\mu }\mathrm{m}$ and $p=\mathcal{L}$.

The accordance between the theoretical ($I_{sd}^T$) and experimental ($I_{sd}^E$) source-drain currents can be quantified by means of the standard deviation (σ), given by

$$\sigma =\sqrt{\frac{1}{N}{\displaystyle \sum _{j=1}^N{\left\{I_{sd}^T[V_G(j)]-I_{sd}^E[V_G(j)]\right\}}^2}},$$

(20)

where $V_G(j)=j-51 \mathrm{volts}$ is the j-th analyzed gate voltage and $I_{sd}^E[V_G(j)]$ are digitalized experimental data (cyan spheres in Figure 7) from reference [29] with $N =101$. The resulting σ for graphene ribbons of $\mathcal{L}=1,\hspace{0.33em}2,\hspace{0.33em}3,\hspace{0.33em}4,\hspace{0.33em}5\hspace{0.33em}\mathrm{and}\hspace{0.33em}6\hspace{0.33em}\mathsf{\mu }\mathrm{m}$ are respectively 3.4423, 3.0119, 2.5801, 2.7210, 1.9327 and 1.4795 μA.

Note in Figure 7 the asymmetry of $I_{sd}$ values with respect to $V_G =0$, whose magnitude diminishes as the ribbon length increases. This asymmetry is derived from that of the contact-resistance ($R_c$) spectrum in ref. [29], which is probably related to the slight doping of the used graphene ribbon [30]. In fact, the contribution of $R_c$ to $I_{sd}$ diminishes as the resistance of graphene ribbon (R) grows [see Equation (15)], while R in turn increases with the ribbon length. Therefore, the asymmetry of $I_{sd}$ respect to $V_G =0$ should decrease as the ribbon length grows.

4. Conclusions

The correlation between source-drain current and gate voltage in graphene field-effect transistors (GFETs) is investigated by means of an atomic-scale tight-binding model, where mesoscopic graphene ribbons with edge reconstruction defects and transversal dislocations are addressed by an independent dual-channel transformation, which converts armchair-edged graphene ribbons into a set of independent dual channels.

The electronic transport was studied within the Landauer formalism, and a new transfer matrix method has been further developed for each dual channel with nearest- and next-nearest-neighbor interactions, including aperiodically placed dislocations following a dilute Rudin–Shapiro (RS) sequence, which is one of the closest aperiodic arrangements to the random distribution. The Landauer conductance was confirmed by that obtained from the Kubo–Greenwood formula (see Appendix B), while the density of states from the Green’s function has been verified by analytical solutions of Equation (19) for the case without dislocations.

Quantized electrical conductance spectra are observed even in presence of edge reconstruction defects along mesoscopic graphene ribbons without dislocations, whose maximum value corresponds to the number of dual channels, while the multi-step behavior is softened at finite temperatures. In addition, the back gate voltage ($V_G$) creates a shift of the chemical potential in graphene ribbons, which produces a V-shape correlation between the source-drain current ($I_{sd}$) and $V_G$ originated from the V-shape DOS spectrum of graphene around the Dirac point. Finally, the realistic calculation of $I_{sd}$ reveals an excellent agreement between the theoretical prediction from a single set of parameters and multiple experimental data obtained from GFETs of six different lengths [29].

The approach of independent dual-channel plus renormalization method presented in this article can be used to study biosensor devices based on GFETs by considering adsorbed molecules as Fano impurities [34]. This study is currently in process.