Consequences of Kondo exchange on quantum spins

Consequences of Kondo exchange on quantum spins

F. Delgado C. F. Hirjibehedin J. Fernández-Rossier111On leave from Departamento de Física Aplicada, Universidad de Alicante, Spain International Iberian Nanotechnology Laboratory (INL), 4715-330 Braga, Portugal. London Centre for Nanotechnology, University College London (UCL), London WC1H 0AH, UK Department of Physics and Astronomy, UCL, London WC1E 6BT, UK. Department of Chemistry, UCL, London WC1H 0AJ, UK

When individual quantum spins are placed in close proximity to conducting substrates, the localized spin is coupled to the nearby itinerant conduction electrons via Kondo exchange. In the strong coupling limit this can result in the Kondo effect - the formation of a correlated, many body singlet state - and a resulting renormalization of the density of states near the Fermi energy. However, even when Kondo screening does not occur, Kondo exchange can give rise to a wide variety of other phenomena. In addition to the well known renormalization of the factor and the finite spin decoherence and relaxation times, Kondo exchange has recently been found to give rise to a newly discovered effect: the renormalization of the single ion magnetic anisotropy. Here we put these apparently different phenomena on equal footing by treating the effect of Kondo exchange perturbatively. In this formalism, the central quantity is , the product of the density of states at the Fermi energy and the Kondo exchange constant . We show that perturbation theory correctly describes the experimentally observed exchange induced shifts of the single spin excitation energies, demonstrating that Kondo exchange can be used to tune the effective magnetic anisotropy of a single spin.

Kondo exchange, spins, single atom, renormalization
journal: Surface Science

1 Introduction

The development of electron paramagnetic resonance made it possible to study the spin transitions of a variety of spin systems, such as paramagnetic molecules Tinkham_PhD_1954 () and transition metal dopants in insulating hosts Abragam_Bleaney_book_1970 (). This led to the development of a single spin Hamiltonian, where the influence of both the Zeeman effect and magnetic anisotropy determine the energy spectrum and spin selection rules. Interestingly, the same type of Hamiltonian was successfully used to describe the quantum spin tunnelling phenomenon Gatteschi_Sessoli_book_2006 () discovered in magnetic molecules with large spin.

Thanks to the tremendous progress in nano-fabrication and nano-manipulation, it is now possible to produce devices where an individual quantum spin can be probed. A single magnetic molecule can be placed in a nanoscale junction Scott_ACSNano_2010 (); Zyazin_Nanolett_2010 (); Parks_Science_2010 (); Vincent_Klyatskaya_nat_2012 (), on top of a carbon nanotube Ganzhorn_Klyatskaya_acs_2013 (), or on a surface Mannini_Nature_2010 (); Kahle_Deng_nanolett_2011 (). A particularly suitable instrument for studying spin systems at the atomic scale is a scanning tunnelling microscope (STM) because it permits not only probing but also manipulation of the spin of individual magnetic atoms deposited on surfaces Wiesendanger_revmod_2009 (); Brune_Gambardella_sursci_2009 (); Gauyacq_Pierre_psc_2012 (), which thereby takes us closer to the Feynman’s dream of engineering matter at the atomic scale. Interestingly, magnetic adatoms can also be described with the same type of single ion Hamiltonian as magnetic dopants in insulating hosts and single-molecule magnets Hirjibehedin_Lin_Science_2007 (). These systems have attracted significant attention because they represent the ultimate limit of magnetic objects where classical or quantum information can be stored Leuenberger_Loss_nature_2001 (); Delgado_Rossier_prl_2012 ().

Manipulation and readout of the information requires integration of these quantized spins (e.g. magnetic molecules, spin chains, or magnetic atoms) into a device. In the case of quantum spins in contact with a conducting electrode, found in many proposed device geometries Bogani_Wernsdorfer_natmat_2008 (), the question of how exchange interaction with the conduction electrons changes the spin dynamics of the quantized spin naturally arises. In the strong coupling regime, the Kondo effect is known to quench the magnetic moment of the quantum spin. This comes together with a strong renormalization of the states at the Fermi energy, which in STM measurements is revealed as a Fano lineshape in the low bias conductance Madhavan_Chen_1998 (); Ternes_JPCM_2009 ().

More recently, the tunnelling spectra of magnetic adatoms Heinrich_Gupta_science_2004 (); Hirjibehedin_Lutz_Science_2006 (); Hirjibehedin_Lin_Science_2007 (); Otte_Ternes_natphys_2008 (); Loth_Bergmann_natphys_2010 (); Khajetoorians_Chilian_nature_2010 (); Bryant_Spinelli_prl_2013 (); Khajetoorians_Schlenk_prl_2013 (); Miyamachi_Schuh_nature_2013 () and molecules Chen_Fu_prl_2008 (); Tsukahara_Noto_prl_2009 () have been found to display inelastic spin transitions, revealed as magnetic field-dependent steps in the differential conductance (see Fig. 1). Fitting the energies of these steps to an effective spin Hamiltonian provides a quantitative understanding of the magnetic anisotropy Hirjibehedin_Lutz_Science_2006 (); Hirjibehedin_Lin_Science_2007 (); Delgado_Rossier_prb_2010 (); Khajetoorians_Chilian_nature_2010 (); Miyamachi_Schuh_nature_2013 (). The steps in are equivalently peaks in , whose half width at half maximum comes from thermal and instrumental smearing as well as the broadening of the transition due to the finite spin lifetime.

Importantly, Kondo exchange influences the quantum spins even in the absence of Kondo effect, i.e. when no Kondo feature is seen in the conductance spectrum. For instance, because of the Kondo exchange, the single-spin states acquire a finite lifetime Langreth_Wilkins_prb_1972 (); Delgado_Rossier_prb_2010 (). In the case of magnetic adatoms, fast spin relaxation times, of the order of 200 fs, have been estimated from the full width at half maximum of the peaks of Fe atoms on a metal Khajetoorians_Lounis_prl_2011 (), while direct STM measurements of the relaxation times of Fe on top of a CuN substrate, possible using pump and probe techniques Loth_Etzkorn_science_2010 (), has demonstrated lifetimes up to 50 ns.

The Kondo exchange can actually arise from two different physical mechanisms. First, direct ferromagnetic exchange is possible between the itinerant electrons of the surface and the or levels of the atomic spin. This type of exchange is responsible, for instance, for the spin splitting of the conduction -type band in diluted magnetic semiconductors Furdyna_jap_1988 (). Second, if the surface electrons hybridize with the localized or orbitals, the so called kinetic exchange Anderson_prl_1966 () results in an antiferromagnetic Kondo coupling, in the limit where classical charge fluctuations of the atom are frozen. This second mechanism is almost ubiquitous and can coexist with the first, giving rise to a reduced total exchange due to their opposite signs.

In this work, we emphasize the central role of the Kondo exchange coupling in a vast variety of available experimental observations of magnetic adsorbates, and thus, we demonstrate that it is possible to quantify its effects. Table 1 shows a summary of physical quantities associated to the spins of a few magnetic impurities that are modified by the exchange coupling to the conduction electrons. Notice that all of them depends on the product of the electrode density of states at the Fermi level, , and the Kondo exchange coupling . The effect can be classified then according to the order in . To first order it leads to a modification of the effective g factor, an effect akin to the Knight-shift in metals. To second order, it leads to finite decoherence and lifetimes Delgado_Rossier_prb_2010 (); Delgado_Rossier_prl_2012 (); Khajetoorians_Lounis_prl_2011 (); Loth_Etzkorn_science_2010 () or the indirect exchange due to the RKKY interaction Kittel_book_1963 (). In addition to these well known results, the Kondo exchange coupling also leads to another second order effect recently observed in magnetic atoms: the renormalization of the magnetic anisotropy Oberg_Calvo_natnano_2013 (). Perturbation theory breaks down either when is not a small parameter, in the case of ferromagnetic , or below the Kondo temperature Hewson_book_1997 (), , in the case of antiferromagnetic .

Quantity Symbol Equation Reference
g factor Wolf_Loose_physlett_1969 ()
Spin relaxation Delgado_Rossier_prb_2010 ()
Spin decoherence Delgado_Rossier_prl_2012 ()
Indirect exchange F(r) Kittel_book_1963 ()
Exchange shift Oberg_Calvo_natnano_2013 ()
Kondo Temperature Hewson_book_1997 ()
Table 1: Physical quantities associated with the Kondo exchange coupling between a magnetic impurity and conduction electrons spins. All of them are determined by the product , with the substrate density of states at the Fermi level.

2 Theoretical approach

2.1 Hamiltonian model

Our starting point is the Hamiltonian Delgado_Rossier_prb_2010 (); Rossier_prl_2009 (); Fransson_nanolett_2009 ()


where is a single spin Hamiltonian discussed below, and describes the independent electrons of the surface


with () the creation (annihilation) operator of an electron in the surface with momentum , spin and single particle energy . Except in Sec. 3, we consider non-magnetic surfaces where . Finally, describes the local exchange interaction between the surface electron density and the magnetic adatoms:


with the vector of Pauli matrices (with eigenvalues) and the s-d exchange interaction between the local spin and the transport electrons. For simplicity, we will assume that these coupling constants are momentum independent and we shall take the average value on the Fermi surface, i.e., , where is a typical length of the macroscopic electrode and its dimensionality (i.e. can be either an area or a volume). Notice that has dimensions of energy times .

In order to keep the ensuing discussion as general as possible, we consider a generic spin Hamiltonian in Eq. (1), where may describe both the electronic and nuclear spin degree(s) of freedom. For specific calculations we will use a Hamiltonian valid for many magnetic systems on surfaces, including Mn, Co and Fe on CuN/Cu Hirjibehedin_Lin_Science_2007 (); Otte_Ternes_natphys_2008 (), Fe-Pc moleculesTsukahara_Noto_prl_2009 () and Fe clusters Khajetoorians_Baxevanis_science_2013 ()


where the first and second terms correspond to the axial and transverse magnetocrystalline anisotropy respectively and stands for the adatom gyromagnetic factor. This Hamiltonian, which neglects the hyperfine coupling, is adequate for a system with 3 nonequivalent magnetic symmetry axis Hirjibehedin_Lin_Science_2007 (). On a surface the term will be most certainly present, but other possibilities involving and are also possible Miyamachi_Schuh_nature_2013 (). In the following we show the influence of the exchange interaction (3) on the dynamics of the anisotropic spin governed by a generic spin Hamiltonian .

2.2 Calculation methodology

In this article we concentrate on the weak coupling regime where a perturbative treatment of the exchange interaction (3) is valid. This means that the dimensionless constant that controls the strength of the exchange coupling, as described below, with the volumetric density of states of the conduction electrons at the Fermi level, satisfies .

We now review the perturbative theory that permits addressing the influence of the Kondo exchange on the spin dynamics and the energy levels of the spin. The main idea is that we treat the anisotropic spin as an open quantum system coupled, via Kondo exchange, to an electronic reservoir, given by the conduction electrons. In principle both the surface and tip electrons affect the atomic spin. The effect of the tip can be made negligible by decreasing the tunnelling amplitude. Hence, we focus on the effect of the surface electrons, although the generalization to include the tip is straightforward Delgado_Rossier_prb_2010 ().

3 First order perturbation theory

To linear order in the Kondo exchange, the electron gas can influence the spin of the magnetic adatom provided that time reversal symmetry is broken, either spontaneously or by an applied field. When that happens, the average magnetization of the electron gas is nonzero. Quantizing the spin along that axis, which we call , and replacing by its average , where is the Fermi Dirac distribution, one gets that for a momentum independent coupling constant , the Kondo coupling of Eq. (3) reads as


Then, if we introduce the total number of electrons with spin , , we get


Thus, at this rough level of approximation, the spin of the magnetic adatom is coupled to the average spin density of the electron gas. In the presence of an applied magnetic field, simple linear response theory yields the well known Pauli paramagnetism result Ashcroft_Mermin_book_1976 ()


where is the gyromagnetic factor of the surface electrons. We can now re-write the Zeeman term as with the renormalized Landé -factor


Thus, to linear order, the effect of the Kondo exchange is to renormalize the factor Wolf_Loose_physlett_1969 (), an effect that can only be measured in the presence of an applied magnetic field and was first proposed in the context of nuclear magnetic resonance shifts in metals, where it is known as Knight shift Knight_pr_1949 (). This -factor renormalization has been recently detected by STM measurements Zhang_Kahle_natcomm_2013 ().

Figure 1: Main effects of the Kondo coupling on the electronic transport. The inelastic spin-flip transitions are revealed as thermally broadened steps in the [panels a) and c)], and peaks (or dips for negative voltage) in the , panels b) and d). As the Kondo coupling grows ( increases, lower panels), the inelastic step shifts to lower energies and it broadens. The black-dotted lines in panels c) and d) represent the shapes of the and respectively considering only the shift in the transition energy and neglecting the change in the broadenings , Eq. (12), while the new shapes appear in red.

4 Second order perturbation theory

To first order in the Kondo coupling, the quantized spin couples only to the average magnetization. To second order, in contrast, the quantized spin couples to the quantum fluctuations of the electron gas magnetization, which occur through the creation of electron-hole pairs across the Fermi energy. To second order in , this coupling has three main consequences on the quantized spin:

  1. The eigenstates of the quantized spin acquire a finite lifetime .

  2. If the quantized spin is prepared in a coherent superposition of states and , it decays in a time scale .

  3. The transition energy is renormalized due to the Kondo exchange .

Whereas the notions of spin relaxation and spin decoherence are well established theoretically and experimentally, and have been worked out in the context of exchanged coupled quantized spins Delgado_Rossier_prb_2010 (), the notion of a reservoir induced shift is less common and it has been only very recently reported in the context of magnetic adatoms Oberg_Calvo_natnano_2013 ().

4.1 Bloch-Redfield quantum master equation

We now show that the second order perturbation theory is able to account for these three physical phenomena. Formally, this is done using the so called system plus reservoir Bloch-Redfield Cohen_Grynberg_book_1998 () approach, in which the dissipative contribution of a reservoir on the otherwise coherent dynamic evolution of a system is calculated up to second order in their coupling. In so doing, we are assuming that the coupling between the quantum system, i.e., the quantum spins, and the electronic reservoir is small, so that the reservoirs stay in its stationary state at thermal equilibrium, producing a force fluctuating about a zero average value with a short correlation time , much shorter than the typical time scales of the spin system Cohen_Grynberg_book_1998 (). In our case, the system is the quantized spin while the reservoir is given by the conduction electrons and the coupling takes the form of the Kondo exchange Delgado_Palacios_prl_2010 (); Delgado_Rossier_prb_2010 ().

The Bloch-Redfield theory yields the dynamical equation for the reduced density matrix Cohen_Grynberg_book_1998 ():


with the Bloch-Redfield tensor, which is a quadratic functional of the system-reservoir coupling and is responsible of the dissipative effects. Here we have employed the secular approximation for the master equation, which basically consist in neglecting the coupling between coherences with very different Bohr frequencies Cohen_Grynberg_book_1998 (). Importantly, in a time scale much longer than the decoherence time , the dynamics of the diagonal terms, , which describe the occupations of the eigenstates of , and off-diagonal terms, , that describe coherences between levels and , are decoupled. The equation for the occupations yields the standard master equation:


where the transition rates from state to , denoted by , are related to for and .

The Bloch-Redfield equation (9) couples coherences to  Cohen_Grynberg_book_1998 () only if the transition energy is degenerate with . In the two specific cases considered here, there is no coupling between different degenerate coherences, so that their equation of motion reads:


Thus, in an isolated system , Eq. (11) describes the evolution of the coherence between two levels and as an oscillating function with angular frequency . The coupling to the reservoir has then two effects on the evolution of the coherences, given by the real and imaginary parts of the Redfield tensor,  Cohen_Grynberg_book_1998 (). First, over a time scale it induces a decay of the amplitude of the oscillation, known as decoherence. The decoherence rate, , has both an inelastic population scattering term, and the pure dephasing rate, , which does not require population scattering Cohen_Grynberg_book_1998 (). Second, it modifies the oscillation frequency , i.e. it induces a shift of the transition energy. Therefore, decoherence and energy shift are the real and imaginary part of the same Bloch-Redfield tensor and are both consequences of the dissipative coupling of a quantum system to a fluctuating reservoir.

In the following we provide explicit expression for the scattering rates, decoherence rates and transition energy shifts for the case of a quantized spin exchanged coupled to an electron gas.

4.2 Transition rates

We consider the simple case where the quantized spin is coupled to a single electronic reservoir that is not spin polarized. The rates in the simpler case read:


where the and denotes the imaginary part of:


with the Fermi function and the electronic density of states. The cases of a spin polarized reservoir and coupling to two reservoirs yield analogous expressions and have been discussed elsewhere Delgado_Palacios_prl_2010 (); Delgado_Rossier_prb_2010 ().

We can give a closed analytical expression for the transition rates, in terms of the spin matrix elements, the Kondo exchange, and the density of states of the conduction electrons at the Fermi energy if we assume a flat density of states with an energy bandwidth , and we neglect the momentum dependence of Kondo exchange . With those assumptions, and taking into account the distribution relation where stands for the Cauchy principal part, Eqs. (12-13) take the form




and . In the limit we can approximate which implies that the spin relaxation rate from to is proportional to the energy released in the transition. In contrast, the same equation yields that uphill transitions are thermally suppressed by a Boltzmann factor. In the elastic case (), we have , which is the well known Korringa results for spin relaxationKorringa_phys_1950 (). Thus, the spin relaxation rate is governed by the dimensionless parameter , the spin selection rules contained in and the phase-space for scattering described by .

4.3 Decoherence rates

The adiabatic decoherence rate for a coherence between two degenerate states and of a quantized spin exchange coupled to a spin unpolarized electron gas, using the same approximations of momentum-independent and flat density of states , reads:

× ∑_σσ’— ∑_a=x,y,z(τ_σσ’^a⟨n—S_a—n⟩-τ_σ’σ^a⟨m—S_a—m⟩)—^2, (16)

where is the -Pauli matrix. Notice that this adiabatic decoherence occurs via elastic scattering. The adiabatic rate scales linearly with because elastic scattering events require that the conduction electron system has an initial occupied state degenerate with a final empty state. As in the case of the scattering rates, decoherence rates is also proportional to .

4.4 Energy shifts

We now write down the expression for the shift of a transition energy between two non-degenerate eigenstates and of the quantized spin Hamiltonian due to their Kondo coupling to an electron gas:


where Re corresponds to the real part. Notice that the shift of a level has contributions coming from spin-matrix elements connecting to all states . At the same level of approximation used to derive Eqs. (14) and (16), we obtain an expression for the shift of an energy level  Oberg_Calvo_natnano_2013 (); Cohen_Grynberg_book_1998 ()




with the digamma function. This expression is valid provided  Bloomfield_Philip_pr_1967 (), which for metals stands even at room temperature. In the regime we are interested in, where the splittings are much smaller than the bandwidth, Eq. (18) can be approximated by its leading order term in :


where is a shift common to all the energy levels, and therefore, not observable. Thus, if we consider the excitation energy of an anisotropic spin system, the renormalized energy difference will be given to leading order in as

× ∑_n’,a [ — ⟨n—S_a—n’⟩—^2Δ_nn’-— ⟨m—S_a—n’⟩—^2Δ_mn’]. (21)

Thus, the renormalization of the transition energy is the difference in the shifts of the levels and , both described with Eq. (17), see Fig. 2a.

4.4.1 Second order correction of the factor for

We first apply Eq. (21) to the case of a spin interacting with a magnetic field. Including the term linear in from Eq. (8), we obtain the following expression up to order :


In the derivation of the contribution quadratic in () to this equation we have ignored the small difference in density of states for different spin orientations, that plays a role in the derivation of the rates Delgado_Rossier_prb_2010 (). By so doing, though, we recover the same expression that was derived using the Kadanoff-Baym Green function method by Langreth and Wilkins Langreth_Wilkins_prb_1972 ().

4.4.2 Shifts for half-integer spins

We now compute the shift of the spin transition for a system with finite spin excitations at zero field, namely, a spin system described with Hamiltonian (4), whose energy levels are shown in figure 2(b).. This, for instance, describes a Cobalt adatom on CuOtte_Ternes_natphys_2008 (); Oberg_Calvo_natnano_2013 () . In that case there is a single transition at zero-field and, for in Eq. (4), the only excitation energy is given by Oberg_Calvo_natnano_2013 ()


where and (see Fig. 2b). In particular, we have that to lowest order in , . The renormalization of the excitation energy has been recently measuredOberg_Calvo_natnano_2013 () for Co adatoms on a CuN substrate, where the presence of a Kondo peak in the conductance permits calibrating the intensity of the exchange coupling. There, the variations of the Kondo coupling throughout the CuN islands led to variations of the magnetic anisotropy by a factor 2, from meV and axial and transversal magnetic anisotropies meV and meV, respectively, to a reduced excitation energy meV and meV and when .

Figure 2: a) Sketch of the renormalization of the energy levels of an anisotropic spin system. b) Modification of the spin levels of a spin system with easy axis anisotropy (). The finite exchange with the substrate electrons induces a reduction of the excitation energy . For finite , each energy level is shifted with a displacement proportional to , leading to an excitation energy . c) Quenching of the zero field splitting of a spin system with the exchange coupling .

4.4.3 Shifts for integer spins

We now apply apply the theory to study the renormalization of the zero-field splitting due to the quantum tunnelling of magnetization present in integer spins when . For simplicity, we consider the example of a spin with easy axis anisotropy () (see figure 2(c)).. The eigenvalues of this system are , and . We assume so that . Using the general expressions for the shifts, Eq. (21), one gets that


where is the bare energy splitting and we have taking into account that the contribution coming from the matrix elements within the doublet is twice the one coming from their coupling to the level, see Eq. (21).

Hence, in the case of integer spins, the Kondo coupling is the responsible for the renormalization of the quantum tunnelling splitting, enabling in this way the decoherence between the two quantum mechanical superposition states and being ultimately responsible of the emergence of the classical magnetic states Delgado_Loth_prep ().

5 Discussion and conclusions

We have reviewed the effect of the Kondo exchange on the spin dynamics of a quantized spin in the weak coupling limit where perturbation theory works. We have discussed four different effects:

  1. The renormalization of the factor, related to the so called Knight shift in nuclear physics (Eq. (8)). This might account in part for the observed anomalously large factor of single Fe atoms adsorbed on a Ag(111) Chilian_Khajetoorians_prb_2011 ().

  2. The finite lifetime of excited spin states, which gives rise to a relaxation rate of excited spin states (Eq. (14)). The linear relation between the rate and the transition energy might account for the observations of for Fe on Ag(111) Chilian_Khajetoorians_prb_2011 () as well as for Fe on Cu(111) Khajetoorians_Lounis_prl_2011 ().

  3. The decoherence of degenerate eigenstates of the spin Hamiltonian [Eq. (16)]. In the case of semi-integer spins with this mechanism ensures that coherence between the two ground states with opposite disappears on a timescale of picoseconds Delgado_Rossier_prl_2012 (), preventing the formation of Schrödinger-cat like states with null magnetization Delgado_Loth_prep ().

  4. The renormalization of the excitation energy [Eq. (21)] that accounts for the recent observation for Co atoms on CuN/Cu(001) Oberg_Calvo_natnano_2013 ().

To this list of physical phenomena, controlled by , that involve quantized spins exchanged coupled to an electron gas, one should of course add the Kondo effect and, when two or more quantized spins are coupled to the same electron gas, the indirect exchange interaction .

In this work we have reviewed the case of a quantized spin couple to a single spin unpolarized electrode (except during the discussion of linear order effects). It is straightforward to extend the theory in two directions. First, one can include a second electrode at a different chemical potential to model inelastic electron tunnel spectroscopy Rossier_prl_2009 (). In this framework, the inelastic current is proportional to , where are the density of states at the Fermi energy of tip and surface and is the Kondo exchange coupling for processes in which the electron tunnels between tip and sample.

The second extension is to consider a spin-polarized electrode. This permits modelling Delgado_Palacios_prl_2010 () two additional effects that have been reported in the literature of magnetic adatomsLoth_Bergmann_natphys_2010 (); Khajetoorians_Lounis_prl_2011 (); Khajetoorians_Wiebe_science_2011 (). For a spin polarized STM tip, the linear conductance depends on the relative orientation of tip and magnetic adatom magnetizations. The spin contrast is linearly proportional to . In addition, spin-polarized currents can control the orientation of the magnetic adatomLoth_Bergmann_natphys_2010 ().

As a final remark, we have to note that whereas the theory presented here looks different from other theory work addressing the same problem Lorente_Gauyacq_prl_2009 (); Khajetoorians_Lounis_prl_2011 (), the underlying physical phenomena are the same. The main advantages of the approach reviewed here are the following. First, it permits connecting the physical phenomena observed in magnetic adatoms with well established effects, proposed in other contexts, such as the Knight shift Knight_pr_1949 () or the Korringa spin relaxation Korringa_phys_1950 (). Second, it identifies a single dimensionless quantity, as the essential parameter that controls the magnitude of the influence of Kondo exchange on the spin dynamics of magnetic adatoms. Third, it connects with a vast body of literature using the Kondo model Wolf_Loose_physlett_1969 (); Langreth_Wilkins_prb_1972 (); Hewson_book_1997 ().


We acknowledge J. C. Oberg, M. R. Calvo, D. Jacob, D. Serrate and M. Moro-Lagares for fruitful discussions. This work was supported by the Engineering and Physical Sciences Research Council UK (EP/D063604/1 and EP/H002367/1); the Leverhulme Trust (RPG-2012-754); Ministry of Science and Education Spain (FIS2010-21883-C02-01, MAT2010-19236, CONSOLIDER CSD2007-0010 and Programa de Movilidad Postdoctoral); European Commission FP7 Programme (PER-GA-2009-251791) and GV grant Prometeo 2012-11.



  • (1) M. Tinkham, Theory of the fine structure of the molecular oxygen ground state with an experimental study of its microwave paramagnetic spectrum, Ph.D. thesis, Massachusetts Institute of Technology (1954).
  • (2) A. Abragam, B. Bleaney, Electron Paramagnetic Resonance of Transition Ions, Oxford University Press, Oxford, 1970.
  • (3) D. Gatteschi, R. Sessoli, J. Villain, Molecular nanomagnets, Oxford University Press, New York, 2006.
  • (4) G. D. Scott, D. Natelson, ACS Nano 4 (2010) 3560.
  • (5) A. S. Zyazin, J. W. G. van den Berg, E. A. Osorio, H. S. J. van der Zant, N. P. Konstantinidis, M. Leijnse, M. R. Wegewijs, F. May, W. Hofstetter, C. Danieli, A. Cornia, Nano Lett. 10 (2010) 3307.
  • (6) J. J. Parks, A. R. Champagne, T. A. Costi, W. W. Shum, A. N. Pasupathy, E. Neuscamman, S. Flores-Torres, P. S. Cornaglia, A. A. Aligia, C. A. Balseiro, G. K.-L. Chan, H. D. Abruna, D. C. Ralph, Science 328 (2010) 1370.
  • (7) R. Vincent, S. Klyatskaya, M. Ruben, W. Wernsdorfer, F. Balestro, Nature 488 (7411) (2012) 357.
  • (8) M. Ganzhorn, S. Klyatskaya, M. Ruben, W. Wernsdorfer, ACS nano 7 (7) (2013) 6225.
  • (9) M. Mannini, F. Pineider, C. Danieli, F. Totti, L. Sorace, P. Sainctavit, M.-A. Arrio, E. Otero, L. Joly, J. C. Cezar, A. Cornia, R. Sessoli, Nature 468 (2010) 417.
  • (10) S. Kahle, Z. Deng, N. Malinowski, C. Tonnoir, A. Forment-Aliaga, N. Thontasen, G. Rinke, D. Le, V. Turkowski, T. S. Rahman, et al., Nano letters 12 (1) (2011) 518.
  • (11) R. Wiesendanger, Rev. Mod. Phys. 81 (2009) 1495.
  • (12) H. Brune, P. Gambardella, Surface Science 603 (10-12) (2009) 1812.
  • (13) J.-P. Gauyacq, N. Lorente, F. D. Novaes, Progress in Surface Science 87 (5) (2012) 63.
  • (14) C. Hirjibehedin, C.-Y. Lin, A. Otte, M. Ternes, C. P. Lutz, B. A. Jones, A. J. Heinrich, Science 317 (2007) 1199.
  • (15) M. N. Leuenberger, D. Loss, Nature 410 (2001) 789.
  • (16) F. Delgado, J. Fernández-Rossier, Phys. Rev. Lett. 108 (2012) 196602.
  • (17) L. Bogani, W. Wernsdorfer, Nature Materials 7 (2008) 179.
  • (18) V. Madhavan, W. Chen, T. Jamneala, M. Crommie, N. Wingreen, Science 280 (5363) (1998) 567.
  • (19) M. Ternes, A. J. Heinrich, W.-D. Schneider, J. Phys.: Condens. Matter 21 (2009) 053001.
  • (20) A. J. Heinrich, J. A. Gupta, C. P. Lutz, D. M. Eigler, Science 306 (2004) 466.
  • (21) C. F. Hirjibehedin, C. P. Lutz, A. J. Heinrich, Science 312 (2006) 1021.
  • (22) A. F. Otte, M. Ternes, K. von Bergmann, S. Loth, H. Brune, C. P. Lutz, C. F. Hirjibehedin, A. J. Heinrich, Nature Physics 4 (2008) 847.
  • (23) S. Loth, K. von Bergmann, M. Ternes, A. F. Otte, C. P. Lutz, A. J. Heinrich, Nature Physics 6 (2010) 340.
  • (24) A. A. Khajetoorians, B. Chilian, J. Wiebe, S. Schuwalow, F. Lechermann, R. Wiesendanger, Nature 467 (2010) 1084.
  • (25) B. Bryant, A. Spinelli, J. J. T. Wagenaar, M. Gerrits, A. F. Otte, Phys. Rev. Lett. 111 (2013) 127203.
  • (26) A. A. Khajetoorians, T. Schlenk, B. Schweflinghaus, M. dos Santos Dias, M. Steinbrecher, M. Bouhassoune, S. Lounis, J. Wiebe, R. Wiesendanger, Phys. Rev. Lett. 111 (2013) 157204.
  • (27) T. Miyamachi, T. Schuh, T. Märkl, C. Bresch, T. Balashov, A. Stöhr, C. Karlewski, S. André, M. Marthaler, M. Hoffmann, et al., Nature 503 (7475) (2013) 242.
  • (28) X. Chen, Y.-S. Fu, S.-H. Ji, T. Zhang, P. Cheng, X.-C. Ma, X.-L. Zou, W.-H. Duan, J.-F. Jia, Q.-K. Xue, Phys. Rev. Lett. 101 (2008) 197208.
  • (29) N. Tsukahara, K. Noto, M. Ohara, S. Shiraki, N. Takagi, Y. Takata, J. Miyawaki, M. Taguchi, A. Chainani, S. Shin, M. Kawai, Phys. Rev. Lett. 102 (2009) 167203.
  • (30) F. Delgado, J. Fernández-Rossier, Phys. Rev. B 82 (13) (2010) 134414.
  • (31) D. C. Langreth, J. W. Wilkins, Phys. Rev. B 6 (1972) 3189.
  • (32) A. A. Khajetoorians, S. Lounis, B. Chilian, A. T. Costa, L. Zhou, D. L. Mills, J. Wiebe, R. Wiesendanger, Phys. Rev. Lett. 106 (2011) 037205.
  • (33) S. Loth, M. Etzkorn, C. P. Lutz, D. M. Eigler, A. J. Heinrich, Science 329 (5999) (2010) 1628.
  • (34) J. K. Furdyna, Journal of Applied Physics 64 (4) (1988) R29.
  • (35) P. W. Anderson, Phys. Rev. Lett. 17 (1966) 95.
  • (36) C. Kittel, C.-Y. Fong, Quantum theory of solids, Vol. 24, Wiley New York, 1963.
  • (37) J. C. Oberg, M. R. Calvo, F. Delgado, M. Moro-Lagares, D. Serrate, D. Jacob, J. Fernández-Rossier, C. F. Hirjibehedin, Nature Nanotechnology 9 (2014) 64.
  • (38) A. C. Hewson, The Kondo Problem to Heavy Fermions, Cambridge University Press, Cambridge, UK, 1997.
  • (39) E. Wolf, D. Losee, Physics Letters A 29 (6) (1969) 334.
  • (40) J. Fernández-Rossier, Phys. Rev. Lett. 102 (2009) 256802.
  • (41) J. Fransson, Nano Lett. 9 (2009) 2414.
  • (42) A. A. Khajetoorians, B. Baxevanis, C. Hübner, T. Schlenk, S. Krause, T. O. Wehling, S. Lounis, A. Lichtenstein, D. Pfannkuche, J. Wiebe, et al., Science 339 (6115) (2013) 55.
  • (43) N. W. Ashcroft, N. D.Mermin, Solid State Physics, Thomson Learning, 1976.
  • (44) W. D. Knight, Phys. Rev. 76 (1949) 1259.
  • (45) Y.-h. Zhang, S. Kahle, T. Herden, C. Stroh, M. Mayor, U. Schlickum, M. Ternes, P. Wahl, K. Kern, Nature communications 4 (2013) 2110.
  • (46) C. Cohen-Tannoudji, G. Grynberg, J. Dupont-Roc, Atom-Photon Interactions, Wiley and Sons, INC., New York, 1998.
  • (47) F. Delgado, J. J. Palacios, J. Fernández-Rossier, Phys. Rev. Lett. 104 (2010) 026601.
  • (48) J. Korringa, Physica 16 (7) (1950) 601.
  • (49) P. E. Bloomfield, D. R. Hamann, Phys. Rev. 164 (1967) 856.
  • (50) F. Delgado, S. Loth, M. Zielinski, J. Fernández-Rossier, in preparation.
  • (51) B. Chilian, A. A. Khajetoorians, S. Lounis, A. T. Costa, D. L. Mills, J. Wiebe, R. Wiesendanger, Phys. Rev. B 84 (2011) 212401.
  • (52) A. Khajetoorians, J. Wiebe, B. Chilian, R. Wiesendanger, Science 332 (6033) (2011) 1062.
  • (53) N. Lorente, J.-P. Gauyacq, Phys. Rev. Lett. 103 (2009) 176601.
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