International
Tables for Crystallography Volume I Xray absorption spectroscopy and related techniques Edited by C. T. Chantler, F. Boscherini and B. Bunker 
Open access
International Tables for Crystallography (2022). Vol. I. Early view chapter
https://doi.org/10.1107/S1574870722001628 Magnetic ordering and its influence on Xray spectroscopies^{a}Diamond Light Source, Harwell Science and Innovation Campus, Didcot OX11 0DE, United Kingdom,^{b}Departament de Física de la Matèria Condensada, Universitat de Barcelona, Martí i Franquès 1, 08028 Barcelona, Spain, and ^{c}Institut de Nanociència i Nanotecnologia, 08193 Barcelona, Spain Xray absorption (XA) spectroscopy enables us to probe the electronic structure and magnetic ordering in, for example, thinfilm systems. The photon–matter interaction contains both nonresonant and resonant terms, but only the latter have a strong sensitivity to the spin and orbital moments of the valence shell. Selection rules in XA provide us with a probe to study the local magnetic ground state. The branching ratio of the spin–orbit split corelevel spectra is proportional to the groundstate spin–orbit interaction and can also provide a measure of the spin state. The angular dependence of the Xray magnetic circular dichroism (XMCD) can be described as a sum over an isotropic and an anisotropic contribution, where the latter is linearly proportional to the axial distortion due to strain. The anisotropic properties of magnetic materials are essential to maintain the preferred magnetization direction. These properties, such as the magnetocrystalline anisotropy energy (MAE), have their origin in the orbital moment anisotropy, which can be studied elementspecifically using angulardependent XMCD. Alternatively, the MAE can also be studied using Xray magnetic linear dichroism (XMLD). Keywords: magnetism; branching ratio; angular dependence; magnetocrystalline anisotropy energy. 
Much progress has been made since the mid1980s in the study of magnetic materials using Xray spectroscopy, an area of research that had previously been the sole domain of neutron scattering. The realization that resonant transitions into the unoccupied valence shell in polarized Xray absorption and scattering experiments can provide unique elementspecific spin and orbital moment information has led to an upturn in theoretical and experimental studies. In this chapter and the next, we will outline some of the many opportunities of magnetic Xray spectroscopies. In order to fully appreciate the underlying principles we introduce the interaction of photons with matter, as well as resonant processes. The isotropic (i.e. nonpolarized) spectrum gives information about the charge distribution and spin–orbit interaction, but the spin and orbital properties can only properly be probed using circularly polarized Xrays.
Many contemporary and future applications of magnetic materials are linked to their anisotropic magnetic properties, such as the magnetocrystalline anisotropy energy (MAE), perpendicular magnetic anisotropy and interfacial magnetic coupling, which have their origin in the spin–orbit interaction (van der Laan, 1998a). It will be shown how the resulting anisotropy in the orbital moment can be probed elementspecifically using the angular dependence of the Xray magnetic circulardichroism (XMCD) signal.
In the relativistic photon–matter interaction Hamiltonian, , the leading terms, which explicitly contain the vector potential A, are (Blume, 1985) where r_{n} and p_{n} are the position vector and momentum operator of the nth electron, respectively, k is the photon wavevector, e is the elementary charge, m is the electron rest mass and c is the speed of light. The first two terms arise from expansion of the kinetic energy operator (1/2m)[p − (e/c)A]^{2}, while the third term comes from the Dirac equation, where σ_{n} is the spinvector operator whose components are the Pauli matrices. For brevity, we will omit the summation over n in the following.
The A · p term in gives the Xray absorption (XA), resonant elastic Xray scattering (REXS) and resonant inelastic scattering (RIXS). The A^{2} term gives, apart from the familiar Thomson scattering, the nonresonant inelastic scattering (NIXS) and Compton scattering. The σ · ∇ × A = σ · B term gives the magnetic scattering.
Converting the matrix element to the length form using the equation of motion where is the groundstate Hamiltonian, and expanding the vector potential where ɛ(k) is the photon polarization vector, gives
The lowest order term is the electric dipole transition operator ɛ · r, which can be written in normalized spherical harmonics as where q = −1, 0, +1 correspond to leftcircular, zlinear and rightcircular photon polarization, respectively.
The electron excited from a core level probes the local unoccupied density of states (DOS). The spectral intensity for qpolarized light is given by Fermi's golden rule, in the case of the electric dipole approximation, as In the presence of a magnetic field the j level is split into m sublevels, and spin–orbit interaction couples the orbital states to the magnetic field. If all directions in space are equivalent, then the atom will be in any of the m levels with equal probability. Therefore, a degenerate, filled state has spherical symmetry, without any spatial orientation. When the symmetry is broken, the state splits into levels with different angular distributions and hence a different polarization dependence. Thus, the energy splitting (i.e. symmetry breaking) and the angular or polarization dependence are two different sides of the same coin.
The above can be formalized by considering that the direct product of the irreducible representations, Γ, for the initial and final states and the transition operator must contain the total symmetric representation, i.e. Γ[ψ_{f}(j′m′)]* × Γ(1, q) × Γ[ψ_{i}(jm)] = A_{1} + …, which in cylindrical symmetry means that −m′ + q + m = 0. Thus, conservation of angular momentum gives the selection rule Δm = m′ − m = q (= 0, ±1). Hence, from the magnetic ground state m only a limited subset of final states can be reached. This means that the spectrum is a fingerprint of the specific ground state with a high sensitivity to crystalfield splitting, spin–orbit interaction, site symmetry and spin configuration. The polarization dependence makes the absorption sensitive to the groundstate magnetic moment. Even with unpolarized light, only a small number of final states can be reached.
The electric dipole operator in equation (6) has spherical components and , resulting in the spectra in which I_{XMCD} arises from the imaginary offdiagonal matrix elements, which require complex wavefunctions (m ≠ 0), where the timereversal symmetry is broken (Kramers' degeneracy).
By taking linear combinations of the I_{q} spectra, the spectral intensity in equation (6) can be separated into a geometrical part and a physical (or dynamic) part, where the latter gives the fundamental spectra
Linearly polarized Xrays measure the charge anisotropy and hence give orientational sensitivity (searchlight effect). While circular polarized light can measure the direction of the magnetic moment, 〈M〉, the XMLD is proportional to 〈M^{2}〉, which apart from ferromagnets and ferrimagnets can also be used for antiferromagnets, which have no net total magnetic moment.
In the XA measurements the signal is averaged over the probed sample volume. This differs from resonant elastic Xray scattering (REXS), where the interference between the scattered photon paths gives information on the longrange structural order and, by using polarized light, also the magnetic order. However, in inelastic scattering, such as NIXS and RIXS, the coherence between the scattered photons is lost.
From equation (6) it can be seen that photons only interact with the orbital part of the wavefunction, whereas the spin moment is conserved in the transition. This orbital sensitivity allows the spin and orbital properties of the ground state to be separated, which enables us to study specific orbital effects such as orbital ordering and the Jahn–Teller effect. Using the sum rules (Thole et al., 1992; Carra et al., 1993), the integrated intensities over the spin–orbit splitcore manifold give the expectation values of the spin and orbital moments in the ground state.
Itinerant models for the electronic structure calculation are based on singleparticle transitions into the empty DOS. Most ab initio methods to calculate the DOS use densityfunctional theory (DFT) plus a meanfield approximation, and for magnetic materials spindependent potentials and spin–orbit interaction have to be taken into account.
DFT calculations can be performed either in real space using multiple scattering (MS) or in reciprocal space using bandstructure methods. The ground state in DFT is expressed as a function of the electron density. Its practical application is called the local (spin) densityfunctional approach (LDA), where the kinetic, nuclear and Hartree potentials are taken into account, with the exchange and correlation effects described by a combined potential. Singleparticle calculations (DFT and LDA) give usually good results for the K edges; however, multiplet calculations are needed for transitionmetal L and M edges and lanthanide and actinide L, M, N and O edges.
Due to the strong corehole interaction in localized materials, the nearedge spectral structure does not display the undistorted unoccupied DOS. The corehole screening contains a monopole and an angular part. While the direct core–valence Coulomb interaction (i.e. the corehole potential) is well screened in molecules and solids, the higherorder terms (the Slater integrals) are poorly screened, causing a multiplet structure. In this case, a singleparticle model will fail and multiplet theory is instead required, which includes the atomic Coulomb and exchange interactions.
The multiplet structure provides a fingerprint for the local ground state, and subtle changes in the magnetic interactions, such as those induced by exchange interaction and spin–orbit interaction, can be distinguished. In the dipole approximation the nearedge spectrum corresponds to resonant transitions, such as d^{n} + ℏω_{i} → p^{5}d^{n+1} in d metals or f^{n} + ℏω_{i} → d^{9}f^{n+1} in f metals. Spectral differences are particularly pronounced when the symmetry of the ground state changes. Crystal and ligandfield interactions can be included in the multiplet code using group theory. Hybridization and chargetransfer interactions can be taken into account using a model Hamiltonian, similar to the Hubbard–Anderson impurity model.
Consider a core level with nonzero orbital quantum number (l_{c} ≠ 0), which is split by spin–orbit interaction into two levels j = l_{c} ± s. The j levels are split into sublevels m_{j} due to core–valence exchange interaction, or in the case of a oneelectron model an effective field acting on the core level. The core p to valence d transitions in the L_{2,3} XA can be described using sum rules and moment analysis. The influence of the groundstate moments on the isotropic spectrum is illustrated in Fig. 1 using the oneelectron model in an itinerant d metal, under the assumption that j is a good quantum number (van der Laan, 1997). The intensity is proportional to the number of d holes, n_{h}, giving an integrated signal with statistical ratio L_{3}:L_{2} = 2:1. The groundstate spin–orbit interaction, 〈l · s〉, shifts spectral weight from the L_{2} to the L_{3} edge. For all other groundstate moment contributions the integrated intensity over the separate L_{3} and L_{2} edges is zero. The orbital moment L_{z}, the spin moment S_{z} and the magnetic dipole term T_{z} = shift the spectral weight to lower energy within the L_{3} peak, causing an asymmetric line shape. In the L_{2} peak the intensity shift is opposite for L_{z}. The charge quadrupole moment Q_{zz} only affects the L_{3} edge. The influence of the spin–orbit interaction is discussed in more detail in Section 6.2.
The most distinctive feature in the isotropic XA spectra is the branching ratio B, which is defined as the fraction of the total transition probability in the 2p_{3/2} manifold. For dmetal L_{2,3} edges, the spin–orbit sum rule can be formulated as (Thole & van der Laan, 1988) Hence, B is proportional to the groundstate expectation value of the angular part of the spin–orbit interaction 〈l · s〉 per d hole. Without valenceband spin–orbit interaction B = ⅔, which represents the statistical ratio. When the initialstate crystalfield term is split into sublevels by a spin–orbit interaction that is small compared with the crystal field, each sublevel has a different branching ratio, decreasing with increasing energy.
If the p_{3/2} and p_{1/2} manifolds are mixed due to electrostatic core–valence interaction, the corelevel angular momentum j is no longer a good quantum number. Highspin states will then have a larger branching ratio on average than lowspin states. Due to the selection rule ΔS = 0 in combination with conservation of angular momentum, a ground state with a higher spin state is then favoured by a transition from a higher corelevel j state (Thole & van der Laan, 1988).
The magnetic anisotropic properties of materials can be studied microscopically and elementspecifically using XMCD, which also allows the spin and orbital contributions to the magnetic moment to be separated.
The angulardependent XMCD can be expressed as a sum over terms that are the product of an energydependent spectrum and an angular distribution. Each of these terms must be invariant under all symmetry operations for the site, i.e. total symmetric. Since the photon polarization is a vector, there can be no more than three different fundamental XMCD spectra in arbitrary symmetry. For orthorhombic lattice symmetry, for example, any XMCD spectrum can be written as the linear combination, where P = −i(ɛ* × ɛ) is the helicity vector, is the sample magnetization and I_{x}, I_{y} and I_{z} are the XMCD spectra for along , and , respectively (van der Laan, 1998b). This means that each XMCD spectrum has a distinct angular dependence, as determined by symmetry.
In axial symmetry I_{y} = I_{x}, and the number of distinct XMCD spectra reduces to two. For small distortions, I_{z} will be similar to I_{x}, which means that it is advantageous to introduce the isotropic and anisotropic (or quadrupolar) XMCD spectra, I_{0} = ⅓(I_{x} + I_{y} + I_{z}) and I_{2} = ⅔I_{z} − ⅓(I_{x} + I_{y}), respectively, which have different shapes and I_{2} ≪ I_{0}. The angulardependent XMCD can be rewritten as where γ and μ are the angles of P and , respectively, with the axis of the axial symmetry, which is usually the sample surface normal. Equation (11) means that the pure I_{0} and I_{2} spectra can be measured in selected geometries using For γ = μ = 54.7°, we obtain I_{XMCD} = I_{0}. For γ = 54.7° and γ − μ = 90°, we obtain I_{XMCD} = I_{2}/2^{1/2}.
The ratio I_{2}:I_{0} gives the amount of distortion of the cubic crystal field by the axial field due to, for example, strain as in the case of MnCr_{2}O_{4} films (van der Laan et al., 2010). In the next section we will apply this formalism to determine the magnetocrystalline anisotropy using the sum rules.
The anisotropic magnetic properties, such as the magnetocrystalline anisotropy energy (MAE), easy magnetization direction, magnetostriction and coercivity, all depend on the orbital moment anisotropy, which can be studied elementspecifically using angulardependent XMCD (Stöhr & König, 1995; van der Laan, 1998a). We limit ourselves here to 3d transition metals. In this case, the spin–orbit constant is small (40–80 meV) compared with the 3d band width of a few eV, so that we can use perturbation theory. Assuming that the majority spin band is completely filled, the MAE will be proportional to the difference between the orbital moments along the easy and hard directions (Bruno, 1989), where the orbital moment is largest along the easy direction. This model was corroborated for a gold/cobalt/gold staircase structure, although a proportionality factor was required to scale the anisotropic part (Weller et al., 1995).
The MAE is defined as , where is along the easy direction of magnetization. Sum rules for the electric dipole transition from a core level can measure the orbital moment tensor of the valence shell up to second rank. Therefore, taking a uniaxial symmetry, where the spin S  M makes an angle φ with , the orbital moment L will be written as a secondrank tensor with reduced spherical harmonic = − ½ = and are the isotropic and anisotropic parts of the orbital moment, respectively. Note that from equation (13), 〈L_{z}〉 = 〈L_{i}〉 + 〈L_{a}〉.
Integrating the XMCD spectra in equation (12) and using the orbital sum rule (Thole et al., 1992), where and w_{z} is the measured integrated intensity for , gives the angular dependence for parallel and transverse geometry as (van der Laan, 1998b) where , w_{0} = 〈L_{i}〉 and w_{2} = 〈L_{a}〉. This gives the angle from L to M as For small anisotropy, the maximum in the angle will be near μ = 45° and proportional to w_{2}/w_{0}.
The angular dependence offers two different ways to measure the magnetic anisotropy, namely in parallel and transverse geometry (Dürr & van der Laan, 1997), which are illustrated in Figs. 2(a) and 2(b), respectively.
The angular dependence of the effective spin moment can be written similarly as where give the (isotropic) spin moment S_{z} and the (anisotropic) magnetic dipole term T_{z}, respectively. Note that .
Using the spin sum rule (Carra et al., 1993) we obtain equation (17) again but now with w_{0} = 〈S_{z}〉 and . The angle from T to M is Note that T_{z} ∝ w_{2} has the properties of a traceless Cartesian tensor. The angular dependence of the various moments is given in Table 1.

Instead of measuring the XMCD with the polarization vector and magnetization direction parallel (P  M) along the different crystal directions, the MAE can also be obtained from a single XMCD measurement in transverse geometry (P ⊥ M and not collinear with easy axes; Dürr & van der Laan, 1996). By forcing the electron spins out of the easy direction using an external magnetic field and measuring the perpendicular component of the orbital moment with the polarization vector perpendicular to the magnetization direction it is possible to directly determine the elementspecific easy direction of magnetization (see Fig. 2b; Dürr et al., 1997).
The MAE can also be obtained from XMLD. Sum rules relate the integrated intensities of the sum and the weighted difference of the XMLD over the L_{2,3} edges to the charge quadrupole moment and the anisotropic part of the spin–orbit interaction, respectively (van der Laan, 1999).
In 3d metals H_{soc} = ζλ, where the radial part ζ is scalar (40–80 eV) and the angular part is the operator λ = l · s, and is a small perturbation, so that the MAE can be expressed in terms of the spin–orbit interaction as Hence, the MAE branching ratio of the XMLD is directly proportional to the MAE.
When all d holes have minority spin, , we can retrieve Bruno's formula (Bruno, 1989) from equation (24), When there are also d holes with majority spin, where L changes sign when S is reversed (timereversal symmetry). In principle, 〈L^{↑}〉 − 〈L^{↓}〉 would be accessible from peak asymmetries. However, the orbital sum rule gives the total projected orbital moment .
The angular dependence of the spin–orbit interaction is where The extra term in equation (27), containing the bipolar spherical harmonic arises from the linear dichroism (van der Laan, 1999). Using the XMLD rule (van der Laan, 1999) we obtain the angular dependence of the spin–orbit interaction, which can then be used in equation (24) to obtain the MAE.
The photon–matter interaction contains an A · p term which becomes large near the coretovalence resonances. Selection rules severely curtail the number of allowed transitions, which makes the spectrum a fingerprint for the specific ground state with a high sensitivity to the crystal field, spin–orbit interaction, site symmetry and spin configuration. The polarization dependence makes the absorption sensitive to the groundstate magnetic moment. Even with unpolarized light only a limited number of final states can be reached. The branching ratio of the spin–orbit split corelevel spectra is proportional to the groundstate spin–orbit interaction and can furthermore provide a measure for the spin state.
The polarized Xray absorption signal from a core level to the valence band depends strongly on the directions of the polarized light and the magnetization with respect to the lattice orientation. By including angulardependent effects we can extend the sum rules which relate the integrated signals over the absorption edges to the expectation values of the spin–orbit coupled groundstate multipole moments. The angular dependence allows us to separate groundstate moments which are indistinguishable in a collinear geometry, such as the spin moment and the magnetic dipole term.
References
Blume, M. (1985). J. Appl. Phys. 57, 3615–3618.Google ScholarBruno, P. (1989). Phys. Rev. B, 39, 865–868.Google Scholar
Carra, P., Thole, B. T., Altarelli, M. & Wang, X. (1993). Phys. Rev. Lett. 70, 694–697.Google Scholar
Dürr, H. A., Guo, G. Y., van der Laan, G., Lee, J., Lauhoff, G. & Bland, J. A. C. (1997). Science, 277, 213–215.Google Scholar
Dürr, H. A. & van der Laan, G. (1996). Phys. Rev. B, 54, R760–R763.Google Scholar
Dürr, H. A. & van der Laan, G. (1997). J. Appl. Phys. 81, 5355–5357.Google Scholar
Laan, G. van der (1997). Phys. Rev. B, 55, 8086–8089.Google Scholar
Laan, G. van der (1998a). J. Phys. Condens. Matter, 10, 3239–3253.Google Scholar
Laan, G. van der (1998b). Phys. Rev. B, 57, 5250–5258.Google Scholar
Laan, G. van der (1999). Phys. Rev. Lett. 82, 640–643.Google Scholar
Laan, G. van der, Chopdekar, R. V., Suzuki, Y. & Arenholz, E. (2010). Phys. Rev. Lett. 105, 067405.Google Scholar
Stöhr, J. & König, H. (1995). Phys. Rev. Lett. 75, 3748–3751.Google Scholar
Thole, B. T., Carra, P., Sette, F. & van der Laan, G. (1992). Phys. Rev. Lett. 68, 1943–1946.Google Scholar
Thole, B. T. & van der Laan, G. (1988). Phys. Rev. B, 38, 3158–3171.Google Scholar
Weller, D., Stöhr, J., Nakajima, R., Carl, A., Samant, M. G., Chappert, C., Mégy, R., Beauvillain, P., Veillet, P. & Held, G. A. (1995). Phys. Rev. Lett. 75, 3752–3755.Google Scholar