Tight-Binding Model for Adatoms on Graphene: Analytical Density of States, Spectral Function, and Induced Magnetic Moment

Tight-Binding Model for Adatoms on Graphene: Analytical Density of States, Spectral Function, and Induced Magnetic Moment

N. A. Pike and D. Stroud Department of Physics, The Ohio State University, Columbus, OH 43210
July 26, 2019

In the limit of low adatom concentration, we obtain exact analytic expressions for the local and total density of states (LDOS, TDOS) for a tight-binding model of adatoms on graphene. The model is not limited to nearest-neighbor hopping but can include hopping between carbon atoms at any separation. We also find an analytical expression for the spectral function of an electron of Bloch vector and energy E on the graphene lattice, to first order in the adatom concentration. We treat the electron-electron interaction by including a Hubbard term on the adatom, which we solve within a mean-field approximation. For finite Hubbard , we find the spin-polarized LDOS, TDOS, and spectral function self-consistently. For any choice of parameters of the tight-binding model within mean field theory, we find a critical value of above which a moment develops on the adatom. For most choices of parameters, we find a substantial charge transfer from the adatom to the graphene host.

73.20.At, 73.20.Fz, 73.22.Pr, 75.70.Ak

I Introduction

Graphene is a well known allotrope of carbon in which the carbons bond in a planar configurationwallace (); novoselov2004 (). As a result, the single graphene sheet is effectively two-dimensionalneto2009 (); saito1998 (). Of the four electrons which occupy the outer shell of a carbon atom, three are in orbitals and form in-plane bonds between the nearest-neighbor carbon atoms, while the fourth occupies a orbital. These orbitals form a band of states which is responsible for many of the characteristic electronic properties of grapheneneto2009 (). Among these properties are a zero band gap at the so-called Dirac point, an electronic dispersion relation that, near the Dirac point, is equivalent to that of massless Dirac fermions, and spin-orbit coupling which is believed to be small because of the low atomic number of carbonneto2009 (); saito1998 (). Graphene has a vast number of potential applications, including photo-voltaic cellswang2008 (), ultracapacitorsliu2011 (); stoller2008 (), and spin-transport electronicsyazyev2008 (); tombros (); swartz ().

Recently, a number of researchers have carried out experimental and theoretical investigations into the effects of adatoms and impurities on both the band structure and localized magnetic moments in graphene. Among these are theoretical studies of carbon vacancies in grapheneLehtinen2004 (); Skrypnyk (); Yazyev2007 (), hydrogen atoms on the surface of graphenesofo2012 (), and several other types of disorder in graphenepereira2008 (); wehling (). In several of these cases and in other workwehling (); Yuan2010 (); Rakhmanov12 (), impurity effects have been treated using a tight-binding model for the electronic structure of graphene and impurities, vacancies, or adatoms. These calculations have, however, either been carried out numerically, or in the limit of energies close to the Dirac point, where the graphene density of states can be approximated as linearwehling1 ().

Density-functional calculations for adatoms on graphene have also been carried out. They have shown that the introduction of an adatom bonded to the surface of graphene can lead to a quasi-localized state with an energy near the Fermi energy and that the wave function of this quasi-localized state includes contributions from the orbitals of neighboring carbon atomssofo2012 (); Yazyev2007 (). In some cases it has been found that, even if the introduced defect or adatom is non-magnetic, a localized magnetic moment can form at the defect siteYazyev2007 ().

In this paper, we extend the previous work on graphene with adatoms in two ways. First, we show that the tight-binding model for adatoms on graphene can, in the limit of low concentrations, be solved analytically in the absence of electron-electron interactions. Specifically, we obtain analytical expressions for the local density of states (LDOS) on the adatom, the total density of states (TDOS) of the adatom-graphene system, and the spectral function for an electron with Bloch vector and energy in graphene in the presence of the adatomBena2009 (). All these results are expressed as a function of the graphene density of states, which itself is known analytically for a nearest-neighbor tight binding modelYuan2010 (); Hobson1953 ().

Secondly, we calculate the magnetic properties of the system using the Hubbard model for the electron-electron interaction, which we treat using a standard mean-field approximation. This treatment leads to a transition between a non-magnetic and magnetic state above a critical value of which depends on the parameters of the tight-binding model. In the presence of a finite our model is basically a special case of the well-known Anderson modelanderson1961 (), but with a linear rather than a constant density of states near the Fermi energy. Our results include not only the magnetic moment on the adatom, but also that on the graphene sheet and the charge transfer from the adatom to the sheet, all as functions of the model parameters.

The remainder of the article is arranged as follows: In Sec. II, we describe the model tight-binding Hamiltonian for the graphene-adatom system. We also describe its generalization to include electron-electron interaction on the adatom via a Hubbard term and the mean-field treatment of this term. In Sec. III, we describe the Green’s function method used to analytically calculate the local density of states on the adatom, the total density of states on the graphene lattice in the presence of the adatom, and the spectral function. In Sec. IV, we present numerical results for the local densities of states, total density of states, and the spectral function for the graphene-adatom system. We also give the local densities of states in the presence of a finite Hubbard within mean-field theory, and give the magnetic moment induced by the adatom, as well as the charge transfer from the adatom to the graphene, as a function of the adatom parameters. In Sec. V, we give a concluding discussion.

Ii The Model Hamiltonian

Graphene is composed of two inter-penetrating triangular lattices, which we will label and , and thus two carbon atoms per primitive cell. In the present work, we are interested in a system consisting of a perfect lattice of graphene plus a single adatom, which we will assume has one atomic orbital. We also assume that the adatom lies at the so-called site, above one of the carbon atoms. It has been found, using ab initio electronic structure calculations, that a several species of adatoms, including hydrogen, fluorine, and gold, do occupy a location above one of the carbon atomsnakada (); chan (); ishii ().

Figure 1: (Color Online) Left: graphene crystal structure showing the two interpenetrating lattices labeled as and and the set of nearest neighbor vectors , , and . Right: first Brillouin zone for graphene showing the high symmetry points. This figure is a modified version of one shown in Ref. neto2009 ().

We treat the graphene-adatom system using a tight-binding Hamiltonian that can, in principle, include hopping between any two carbon atoms. For pure graphene, the Hamiltonian can be written in terms of the creation and annihilation operators for electrons of spin on a site in the primitive cell of the and sublattices. We denote the creation (annihilation) operators for the and sublattices by () and (). The corresponding tight-binding Hamiltonian for graphene may be written in real space as


Here and () are hopping integrals which take an electron of spin () from a lattice site to a neighboring lattice site, and denotes a Bravais lattice vector of the triangular lattice. The first sum represents hopping between sublattices and therefore all possible Bravais lattice vectors are summed over, whereas the second sum only includes hopping between sites on the same sublattice and thus, is not allowed. We have assumed that the hopping integrals for hopping on the same sublattice are identical for the and sublattices and therefore set .

Eq. (1) can be Fourier transformed as


where and . In the limit of only nearest neighbor hopping, , and except for the three nearest neighbors. In this limit, we write . The three nearest neighbor vectors are shown in Fig. 1, where they are denoted by , , and . In this limit,


Here the operator , where is the number of primitive cells in the graphene lattice and is the n Bravais lattice vector of the triangular lattice; an analogous definition holds for . The sum over is confined to the first Brillouin zone and is given by Rakhmanov12 ()


In Eq. (4), is the hopping energy between nearest neighbor carbon atoms ( for grapheneRakhmanov12 ()), and is the nearest-neighbor bond lengthYazyev2007 ().

Figure 2: (Color Online) Density of states per spin and per primitive cell for the tight-binding model defined by Eqs. (3) and (4) for the orbitals of graphene, as calculated from (22)Hobson1953 (); Yuan2010 (). Following Ref. Rakhmanov12 (), we assume for graphene.

We wish to investigate what happens to the density of states when when an isolated adatom is adsorbed onto the host graphene at a sitenakada (); chan (). The extra piece of the tight-binding Hamiltonian, , due to the adatom may be written in real space as


Here and are creation and annihilation operators for an electron of spin () at the site of the adatom, which we assume is located at the site of the sublattice, is the on-site energy of an electron on that site (relative to the Dirac point of the pure graphene band structure), and , (), is the energy for an electron to hop between the adatom and the carbon atom at the site of the sub-lattice.

We now wish to express in terms of Bloch eigenstates of . These eigenstates may be written as two-component column vectors with components and satisfying the eigenvalue equation (hereafter we suppress the spin subscript until needed)


The solution to this eigenvalue problem is


which gives the tight-binding band structure of pure grapheneRakhmanov12 (), and the corresponding eigenvectors satisfy


where the phase factor is given by


We can then write the destruction operator for a Bloch electron in the upper band as


and in the lower band as


where we have defined and to be properly normalized, so that, for example, the anticommutator .

With these definitions, we can now use the inverse Fourier transform of the and to obtain


Thus, we can rewrite the impurity Hamiltonian (5) in momentum space as


Thus, in , the creation and annihilation operators of the adatom are connected to every eigenstate of the graphene band structure by matrix elements of equal magnitude (though different phase). For a hydrogen adatom, we take and , as found in Rakhmanov12 (). The one-electron Hamiltonian, , is a special case of the Anderson impurity modelanderson1961 (), where the impurity state is coupled to all the band electron states by matrix elements of equal magnitude.

We also include in our calculation the effects of an on-site electron-electron interaction of the Hubbard form,


where is the number of electrons with spin on the hydrogen site. For a hydrogen adatom we take to be the difference between the ionization potential and the electron infinity providing us with a numberical value of pariser (); lykk ().

The Hubbard term given in Eq. (14) is quartic in the creation and annihilation operators. Therefore, in order to calculate the properties of the Hamiltonian including this term, we use a standard mean field theory to rewrite this term (see, e. g., Ref. Fazekas1999 ()) in the form


With this approximation, the total Hamiltonian, consisting of the sum of Eqs. (3), (13), and (15), becomes quadratic in electron creation and annihilation operators, and can be diagonalized. The Fermi energy, total energy, and magnetic properties of the system can then be obtained by an iterative process as described below. The electronic density of states corresponding to the one-electron Hamiltonian, , can be obtained analytically, as we describe below, which makes the calculation of the total energy and the magnetic properties quite simple.

Iii Green’s function, Density of States, and Spectral Function of Graphene-Adatom System

iii.1 Green’s Function

We use the single particle Green’s function approach to calculate the local and total density of states of the graphene-adatom system, initially omitting the Hubbard-U term. We continue to suppress the spin degree of freedom since, in the absence of the Hubbard term, spin just gives an extra factor of 2. To that end, we first introduce the resolvent operator


where (), and . If there are carbon atoms and 1 adatom, can be expressed as an -dimensional matrix. It is convenient to use the 2N Bloch states (corresponding to values) created by the operators and as the basis for this matrix, plus the adatom orbital corresponding to . If we let the adatom orbital correspond to the first of the states, then one can easily write out the matrix of which is the inverse.

iii.2 Density of States

We denote the local electronic density of states per spin on the adatom site by . is related to by


Here , (), and denotes the matrix element of evaluated at the location of the adatom, which we take to be above the atom on the sub-lattice. This corresponds to an element in the first row and first column of the matrix . We can obtain this matrix element as


where cof denotes the cofactor of the element in the first row and first column of the matrix , and the denominator is the determinant of . Both quantities are readily evaluated, and the result for is




and is given by Eq. (7).

is related to the (unperturbed) graphene density of states per graphene unit cell (per spin), which we denote , by


with anderson1961 (); wehling (). For the form of which includes only nearest neighbor hopping, isHobson1953 (); Yuan2010 ()


where , and is the elliptic integral of the first kind. We plot Eq. (22) in Fig. (2) normalized such that .

is related to Eq. (22) via the principal value integralanderson1961 (); wehling ()


where the integral runs over the range where . The density of states on the carbon sites (per spin) in the presence of an adatom may be written as , where , (). Each of the elements of this sum can be computed using the analog of Eq. (18), with the result


The total density of states per spin is is the sum of the expressions in Eqs. (19) and (24), and can be rearranged to have the form


iii.3 Spectral Function

We can use an analogous approach to calculate the spectral function . represents the probability density that an electron with Bloch wave-vector has energy , and is given by


These matrix elements can be evaluated using the methods of the preceding section, with the result


It is convenient to write this spectral function in terms of a self-energy as


where is readily computed by equating Eqs. (27) and (28). To first order in , is found to be independent of both and and to take the form


All these equations [(19), (20), (21), (23)-(25), (28), and (29)] remain valid for non-nearest-neighbor hopping; only the form of the graphene density of states has to be changed.

iii.4 Effects of Electron-Electron Interaction; Spin-Polarized Density of States and Magnetic Moment

Finally, we discuss the effects of including a non-zero Hubbard term [Eq. (14)] in the Hamiltonian. If we treat by mean-field theory [Eq. (15)], then the densities of states for spin-up and spin-down electrons may be different. We can calculate these partial densities of states self-consistently as follows. First, we make an initial assumption for the value of and . Then the effective on- site energy for an up-spin electron on the hydrogen adatom is obtained by making the replacement


with a corresponding expression for . Given and , we can compute the local densities of states and using the appropriate generalizations of Eq. (19); we can also obtain the total densities of states and using the corresponding generalizations of Eq. (25). The Fermi energy, , is then obtained from the condition


where we assume one adatom, carbon sites, and . Given , we then recalculate and . The procedure is repeated until successive iterations do not lead to a significant change in and . In practice, we require that these quantities change by no more than on successive iterations (here is the number of adatoms in the calculation). Typically, about twenty iterations of the self-consistent equations are needed to attain this degree of convergence, as discussed further below.

Once has been found, the total magnetic moment of the system is obtained from


where is the Bohr magneton.

In the limit , the mean-field version of the Hubbard model can be done without iteration. In this limit, only one of the quantities or is non-zero. The reason is that if, say, is non-zero, then the energy to put a spin-down electron on the adatom becomes infinite, and hence the number of spin-down electrons must be zero. To be definite, we assume that . In that case, we just have , and . The total density of states for the up spins will then be given by Eq. (25), while that for the down spins is just that of unperturbed graphene: .

In the limit the Fermi energy, , is obtained from Eq. (31) and may be simplified to


Once has been obtained, the magnetic moment can be again found using Eq. (32). Since both and are available analytically, using Eqs. (32) and (33), is easily computed in closed form.

Iv Numerical Results

In Fig. 3(a), we plot the local density of states for parameters appropriate to a hydrogen adatom on graphene with , as calculated from Eq. (19). We use the parameters , , and , as given by Ref. Rakhmanov12 () for a hydrogen adatom. In Fig. 3(b), we plot the change in the total density of states produced by a single hydrogen atom, i. e., the quantity for the three cases of Fig. 3(a), calculated using Eqs. (17) and (25).

Next, we calculate both the spectral function for and the spin polarized spectral function for as functions of for several values of , using the parameters of Fig. 2. is obtained using a generalization of Eq. (28) in the limit as discussed in subsection III.4. The resulting spectral functions are shown in Fig. 4 through first order in . The contribution from the adatom appears as the sharp spike near , while the contribution from the graphene sheet is shown as broadened peaks near the values of for the three choices of . The self energy term [Eq. (29)] controls the width of the graphene resonances. The integral of the graphene sheet’s contribution to the spectral function will be of order times larger then that of the adatom. Furthermore, the width of the graphene peaks in the spectral function is proportional to the density of adatoms.

Figure 3: (Color Online) (a). Local density of states per spin on the adatom site, (E), with for a graphene sample with N = 500 graphene unit cells (1000 C atoms) and one adatom. We assume the model described in the text [Eqs. (3), (4), and (13)]. Black curve: , ; blue curve: t, ; and red curve: t, . In all three cases, . The Fermi energy is calculated using Eq. (31) and gives . (b). The change in the density of states per spin due to the adatom for the three cases shown in (a). In both (a) and (b), the insets are enlargements of the region between -1 eV and +1 eV.
Figure 4: (Color Online) (a)-(c). Spectral function at for the graphene-adatom system, as calculated using Eqs. (28) and (29) for three values of corresponding to , , and respectively, assuming a nearest-neighbor tight-binding band. We use , , , and . (d). The spin polarized spectral function for the point and the case in the mean-field approximation, using the same parameters as in (a)-(c). for the majority spin component is shown in black and that of the minority component in red. For the minority spin component, is just that of the unperturbed graphene sheet, i. e., delta functions at the unperturbed pure graphene energy eigenvalues for all values of . For the case , and for the majority spin at , the adatom contribution occurs near , while the graphene sheet contribution corresponds to broadened peaks near the unperturbed energy eigenvalues given in Eq. (7). For points and , the integral of the peak near is of order 1/(2N) times those of the main peaks in the spectral function, and thus vanishes as .
Figure 5: (Color Online) Spin-polarized local density of states (sLDOS) per adatom for both the majority spin (black solid line) and minority spin (red solid line), as obtained by substituting Eq. (30) into Eq. (19). We use and the following values of the on-site energy , hopping energy , and Hubbard energy : (a). ; (b). ; (c) (d). ; (e). ; (f). ; (g). ; (h). .
Figure 6: Total magnetic moment on the adatom and the graphene (), in units of , versus for two values of (Red curve: , Black curve ). In this plot, we hold and as we vary for two different choices of . In both cases, the moment seems to become nonzero at a characteristic value of , which depends on , , and . Lines connect calculated points.

Using the mean-field methods described in section II we can calculate a variety of other spin-independent and spin-dependent properties of the adatom-graphene system. These include and , the local density of states of up and down spin on the adatom; the induced magnetic moment on the adatom () and in the entire system of graphene sheet plus adatom (); and the net charge transfer from the adatom to the sheet, all as functions of the parameters , , and . The magnetic moment on the adatom site is . is obtained from


where () is defined using the appropriate generalization of Eq. (19). The total magnetic moment is given in Eq. (32). The net charge transfer from adatom to the graphene lattice is obtained by first integrating up to the Fermi energy, to obtain the net number of electrons on the adatom, then subtracting this quantity from the adatom valence (i. e., for hydrogen, Z = 1) to obtain the net charge transfer.

We have carried out these calculations for various values of the adatom on-site energy , Hubbard parameter , and hopping energy . In Table I we summarize the results above for parameters appropriate to a hydrogen adatom and summarize the trends when the various adatom parameters are varied. Additional results are shown in Figs. 3 and 5. As can be seen in Table I and Fig. 5, the parameter values thought to be appropriate to an adatom (, , and ), lead to a very small magnetic moment on the adatom though there is an increase in both the LDOS and TDOS close to the Fermi energy (; see Fig. 5(b)).

Summary of Numerical Results
U () Charge
(eV) (eV) per () Transfer (eV)
adatom ()
5.8 0.0 0.372
5.8 2.67E-4 1.13E-3 0.695 0.173
0.4 5.8 3.11E-3 7.67E-3 0.758 0.236
0.300 0.871 0.699 0.111
5.8 0.260 0.927 0.738 0.050
5.8 0.338 0.958 0.662 0.050
5.8 0.360 0.990 0.639 -0.01
0.4 1.8 0.358 0.506 0.641 0.236
0.4 7.8 0.219 -0.11 0.780 0.236
Table 1: Magnetic moment on the adatom (), total magnetic moment on the graphene-adatom system () (both in units of ), and charge transferred from the adatom to the graphene lattice (in units of an electron charge), for various choices of , on-site energy , and hopping energy . Note that , , and corresponds to the expected parameters of a hydrogen adatom. When , we find a spin polarized state near the Fermi energy. The magnetic moment calculated on the adatom is done using a combination of Eqs. (15) and (19) and the magnetic moment on the sheet is calculated using Eq. (32). (a)- Spin polarized LDOS plotted in Fig. (3). (b)- Spin polarized LDOS plotted in Fig. (5b).

In general, as seen in Table I, for sufficiently large , a nonzero magnetic moment develops on both the adatom and the graphene sheet. The moment on the adatom is of order in this limit, for the given parameters, while the sum of the moments on the adatom and the sheet approaches in this limit. We also find in all of our calculations that a large fraction (typically of the electron) is transferred from the adatom to the graphene sheet for the parameters we consider. For the parameters appropriate to hydrogen adatoms, the model predicts no, or only a very small, induced magnetic moment. A possible explanation is that our model assumes no lattice distortion due to the adatom. But DFT calculations have shown that the surface of graphene is warped due to the addition of an adatom. This warping could change the distance between the adatom and the neighboring carbon atoms, and hence possibly the value of the Coulomb integral.

In Fig. 6, we show the total magnetic moment of the system as given by Eq. (32) plotted as a function of , for various values of . In each case shown, and . In all the plots, there is an apparent threshold behavior: the moment becomes nonzero only if exceeds a threshold value which depends on as well as on . While these calculations are done using a simple mean-field approximation, they seem to be consistent with other work on related modelsanderson1961 (); fradkin ().

V Discussion

Using a tight-binding model we have calculated the local and total density of states and the spectral function for a system consisting of a single adatom in a site on graphene. Because the hopping integral from the adatom to a graphene Bloch state has the same magnitude for any , we have shown that these quantities can be calculated analytically. This simplification holds even if we do not make the oft-used linear approximationwehling () for the graphene density of states near the Dirac point. It is also valid even if we include non-nearest-neighbor hopping in the tight-binding graphene Hamiltonian. Since our numerical results give both the local and total density of states, we can compute the charge transfer from the adatom to the graphene. Our numerical results show that, for most parameters we consider, this charge transfer is a substantial fraction of an electron (approximately for parameters appropriate to hydrogen).

Because the calculations are at low adatom concentration, the adatom-induced density of states is linear in concentration. Other work has treated the same system at higher adatom concentration, but only numericallyRakhmanov12 (). In future work, it might be possible to treat the present model analytically at higher concentrations, at least approximately. It would also be of interest to include effects of lattice distortions, which are known to exist when adatoms bind to graphene boukhvalov (), and which can lead to a large increase in spin-orbit interactions neto (); Gmitra (). Such spin-orbit interactions would likely have a large effect on the magnetic properties arising from the adatom.

We have also calculated the magnetic properties induced by the adatom, using a Hubbard model treated within mean-field theory. For all choices of the Hamiltonian parameters, we find that there is a critical value of the Hubbard above which the density of states near the Fermi energy is spin-polarized and a net induced magnetic moment is formed. The appearance of this magnetic moment was predicted long ago to occur within mean-field theory for models with a slowly varying density of states near the Fermi energyanderson1961 (). Here, it is also found to occur in a system with a roughly linear density of states near . While the mean-field approximation is probably unreliable for this model, we note that a similar threshold for moment formation was also found, within the Kondo Hamiltonian, for a system with a linear density of statesfradkin (). Since, at large , it is known that the Hubbard model can be approximately transformed into the Kondo modelschrieffer (), it seems plausible that there could really be a threshold behavior in the Hubbard model with a linear density of state such as is found here, even though we use a mean field theory to obtain it.

A somewhat counterintuitive result of our calculations is that, as increases, the value of needed to induce a magnetic moment becomes smaller. Since a larger suggests that it is easier for the electron to hop from the impurity to the graphene, one might expect that a moment on the impurity atom would be less likely to form. A possible explanation is that the larger also causes the peak in the impurity density of states to shift closer to the Dirac point, where the graphene density of states is smaller. Thus, there are fewer final states available for an electron to hop into, and hence, the electron is less likely to hop, thus increasing the likelihood of moment formation on the impurity.

In our approximation we also calculate the spectral function of our graphene-adatom system to first order in . The main effect of the adatom is, as expected, simply to broaden the delta-function peaks that the spectral function would exhibit in an ideal graphene lattice. In our approach, this broadening, and the shape of the spectral line, are computed analytically. To the same order, we find that both the adatom contribution to the spectral function at and the broadening of the graphene spectral lines will vanish as .

In summary, we have, using a single-particle Green’s function approach together with a tight binding Hamiltonian in the limit of no electron-electron correlations, obtained analytical equations for the LDOS, TDOS, and spectral function for adatoms on the surface of graphene. Using the same model with a finite Hubbard energy , we find that a magnetic moment is induced both on the adatom and nearby on the graphene sheet above a critical value of which depends on the other model parameters. These results are not only of intrinsic interest but also may be useful in understanding the behavior of a variety of adatoms on graphene.

Vi Acknowledgments

This work was supported by the Center for Emerging Materials at The Ohio State University, an NSF MRSEC (Grant No. DMR0820414) . We thank Prof. Roland Kawakami for valuable discussions.


  • (1) P. R. Wallace, Phys. Rev. 71, 662 (1947).
  • (2) K. S. Novoselov, A. K. Geim, S. V. Morozov, D. Jiang, Y. Zhang, S. V. Dubonos, I. V. Grigorieva, and A. A. Firsov, Science 306, 666 (2004).
  • (3) A. H. Castro Neto, F. Guinea, N. M. R. Peres, K. S. Novoselov, and A. K. Geim,  Rev.  Mod.  Phys. 81  109  (2009).
  • (4) R. Saito, G. Dresselhaus, and M. S. Dresselhaus,  Physical Properties of Carbon Nanotubes (Imperial College Press, London, 1998).
  • (5) X. Wang, L. Zhi, and K. Mullen, Nano Letters 8, 323 (2008).
  • (6) W. Liu, T. Dang, Z. Xiao, Z. Li, C. Zhu, and X. Wang, Carbon. 49, 884 (2011).
  • (7) M. D. Stoller, S. Park, Y. Zhu, J. An, and R. Ruoff, Nano Letters 8, 3498 (2008).
  • (8) O. V. Yazyev and M. I. Katsnelson, Phys. Rev. Lett. 100, 047209 (2008).
  • (9) N. Tombros, C. Jozsa, M. Popinciuc, H. T. Jonkman, and B. J. van Wees, Nature 448, 06037 (2007).
  • (10) K. M. McCreary, A. G. Swartz, W. Han, J. Fabian, and R. K. Kawakami, Phys. Rev. Lett. 109, 186604 (2012).
  • (11) P. O. Lehtinen, A. S. Foster, Yuchen Ma, A. V. Krasheninnikov, and R. M. Nieminen. Phys. Rev. Lett. 93, 187202 (2004).
  • (12) O. V. Yazyev and L. Helm, Phys. Rev. B 75, 125408 (2007).
  • (13) Y. V. Skrypnyk and V. M. Loktev, Phys. Rev. B 73, 241402(R) (2006).
  • (14) J. O. Sofo, G. Usaj, P. S. Cornaglia, A. M. Suarez, A.  D. Hernández-Nieves, and C. A. Balseiro. Phys. Rev. B 85, 115405 (2012).
  • (15) V.Ṁ. Pereira, J. M. B. Lopes dos Santos, and A. H. Castro Neto, Phys. Rev. B 77, 115109 (2008).
  • (16) T. O. Wehling, M. I. Katsnelson, and A. I. Lichtenstein, Chem. Phys. Lett. 476 125 (2009).
  • (17) A. L. Rakhmanov,  A. V. Rozhkov, A. O. Sboychakov, and F. Nori. Phys. Rev. B 85, 035408 (2012).
  • (18) S. Yuan, H. De Raedt, and M. I. Katsnelson,  Phys. Rev. B 82, 115448 (2010).
  • (19) T. O. Wehling, A. V. Balatsky, M. I. Katsnelson, A. I. Lichtenstein, K. Scharnberg, and R. Wiesendanger, Phys. Rev. B75, 125425 (2007).
  • (20) C. Bena and G. Montambauz, New J. Phys. 11, 0950003 (2009).
  • (21) J. Hobson and W. A. Nierenberg, Phys. Rev. 86, 662 (1953).
  • (22) P. W. Anderson, Phys. Rev. 124, 41 (1961).
  • (23) K. Nakada and A. Ishii, Solid State Commun. 151, 13 (2011).
  • (24) K. T. Chan, J. B. Neaton, and M. L. Cohen, Phys. Rev. B 77, 235430 (2008).
  • (25) A. Ishii, M. Yamamoto, H. Asano, and K. Fujiwara. J. Phys. Conf. Ser. 100, 052087 (2008).
  • (26) R. Pariser and R. Parr, J. Chem. Phys. 21, 767-775 (1953).
  • (27) K. R. Lykke, K. K. Murray, and W. C. Lineberger, Phys. Rev. A 43, 6104-6107 (1991).
  • (28) P. Fazekas, Lecture Notes on Electron Correlation and Magnetism, (World Scientific, Singapore, 1999).
  • (29) D. W. Boukhvalov, M. I. Katsnelson, and A. I. Lichtenstein, Phys. Rev. B 77, 035427 (2008).
  • (30) A. H. Castro Neto and F. Guinea. Phys. Rev. Lett. 103, 026804 (2009).
  • (31) Martin Gmitra, Denis Kochan, and Jaroslav Fabian, Phys. Rev. Lett. 110 246602 (2013).
  • (32) D. Withoff and E. Fradkin, Phys. Rev. Lett. 64, 1835 (1990).
  • (33) J. R. Schrieffer and P. A. Wolff, Phys. Rev. 149, 491 (1966).
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
Add comment
Loading ...
This is a comment super asjknd jkasnjk adsnkj
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test description