Zeeman effect

The Zeeman effect (/ˈzmən/; Dutch pronunciation: [ˈzeːmɑn]), named after the Dutch physicist Pieter Zeeman, is the effect of splitting of a spectral line into several components in the presence of a static magnetic field. It is analogous to the Stark effect, the splitting of a spectral line into several components in the presence of an electric field. Also similar to the Stark effect, transitions between different components have, in general, different intensities, with some being entirely forbidden (in the dipole approximation), as governed by the selection rules.

Since the distance between the Zeeman sub-levels is a function of magnetic field strength, this effect can be used to measure magnetic field strength, e.g. that of the Sun and other stars or in laboratory plasmas. The Zeeman effect is very important in applications such as nuclear magnetic resonance spectroscopy, electron spin resonance spectroscopy, magnetic resonance imaging (MRI) and Mössbauer spectroscopy. It may also be utilized to improve accuracy in atomic absorption spectroscopy. A theory about the magnetic sense of birds assumes that a protein in the retina is changed due to the Zeeman effect.[1]

When the spectral lines are absorption lines, the effect is called inverse Zeeman effect.


Historically, one distinguishes between the normal and an anomalous Zeeman effect (discovered by Thomas Preston in Dublin, Ireland[2]). The anomalous effect appears on transitions where the net spin of the electrons is an odd half-integer, so that the number of Zeeman sub-levels is even. It was called "anomalous" because the electron spin had not yet been discovered, and so there was no good explanation for it at the time that Zeeman observed the effect.

At higher magnetic field strength the effect ceases to be linear. At even-higher field strength, when the strength of the external field is comparable to the strength of the atom's internal field, electron coupling is disturbed and the spectral lines rearrange. This is called the Paschen-Back effect.

In the modern scientific literature, these terms are rarely used, with a tendency to use just the "Zeeman effect".

Theoretical presentation

The total Hamiltonian of an atom in a magnetic field is

where is the unperturbed Hamiltonian of the atom, and is the perturbation due to the magnetic field:

where is the magnetic moment of the atom. The magnetic moment consists of the electronic and nuclear parts; however, the latter is many orders of magnitude smaller and will be neglected here. Therefore,

where is the Bohr magneton, is the total electronic angular momentum, and is the Landé g-factor. A more accurate approach is to take into account that the operator of the magnetic moment of an electron is a sum of the contributions of the orbital angular momentum and the spin angular momentum , with each multiplied by the appropriate gyromagnetic ratio:

where and (the latter is called the anomalous gyromagnetic ratio; the deviation of the value from 2 is due to the effects of quantum electrodynamics). In the case of the LS coupling, one can sum over all electrons in the atom:

where and are the total orbital momentum and spin of the atom, and averaging is done over a state with a given value of the total angular momentum.

If the interaction term is small (less than the fine structure), it can be treated as a perturbation; this is the Zeeman effect proper. In the Paschen–Back effect, described below, exceeds the LS coupling significantly (but is still small compared to ). In ultra-strong magnetic fields, the magnetic-field interaction may exceed , in which case the atom can no longer exist in its normal meaning, and one talks about Landau levels instead. There are intermediate cases which are more complex than these limit cases.

Weak field (Zeeman effect)

If the spin-orbit interaction dominates over the effect of the external magnetic field, and are not separately conserved, only the total angular momentum is. The spin and orbital angular momentum vectors can be thought of as precessing about the (fixed) total angular momentum vector . The (time-)"averaged" spin vector is then the projection of the spin onto the direction of :

and for the (time-)"averaged" orbital vector:


Using and squaring both sides, we get

and: using and squaring both sides, we get

Combining everything and taking , we obtain the magnetic potential energy of the atom in the applied external magnetic field,

where the quantity in square brackets is the Landé g-factor gJ of the atom ( and ) and is the z-component of the total angular momentum. For a single electron above filled shells and , the Landé g-factor can be simplified into:

Taking to be the perturbation, the Zeeman correction to the energy is

Example: Lyman-alpha transition in hydrogen

The Lyman-alpha transition in hydrogen in the presence of the spin–orbit interaction involves the transitions


In the presence of an external magnetic field, the weak-field Zeeman effect splits the 1S1/2 and 2P1/2 levels into 2 states each () and the 2P3/2 level into 4 states (). The Landé g-factors for the three levels are:

for (j=1/2, l=0)
for (j=1/2, l=1)
for (j=3/2, l=1).

Note in particular that the size of the energy splitting is different for the different orbitals, because the gJ values are different. On the left, fine structure splitting is depicted. This splitting occurs even in the absence of a magnetic field, as it is due to spin-orbit coupling. Depicted on the right is the additional Zeeman splitting, which occurs in the presence of magnetic fields.

Possible transitions for the weak Zeeman effect
Initial state


Initial energy perturbation Final state


Strong field (Paschen–Back effect)

The Paschen–Back effect is the splitting of atomic energy levels in the presence of a strong magnetic field. This occurs when an external magnetic field is sufficiently strong to disrupt the coupling between orbital () and spin () angular momenta. This effect is the strong-field limit of the Zeeman effect. When , the two effects are equivalent. The effect was named after the German physicists Friedrich Paschen and Ernst E. A. Back.[3]

When the magnetic-field perturbation significantly exceeds the spin-orbit interaction, one can safely assume . This allows the expectation values of and to be easily evaluated for a state . The energies are simply

The above may be read as implying that the LS-coupling is completely broken by the external field. However and are still "good" quantum numbers. Together with the selection rules for an electric dipole transition, i.e., this allows to ignore the spin degree of freedom altogether. As a result, only three spectral lines will be visible, corresponding to the selection rule. The splitting is independent of the unperturbed energies and electronic configurations of the levels being considered. In general (if ), these three components are actually groups of several transitions each, due to the residual spin-orbit coupling.

In general, one must now add spin-orbit coupling and relativistic corrections (which are of the same order, known as 'fine structure') as a perturbation to these 'unperturbed' levels. First order perturbation theory with these fine-structure corrections yields the following formula for the Hydrogen atom in the PaschenBack limit:[4]

Possible Lyman-alpha transitions for the strong regime
Initial state


Initial energy Perturbation Final state


Intermediate field for j = 1/2

In the magnetic dipole approximation, the Hamiltonian which includes both the hyperfine and Zeeman interactions is

where is the hyperfine splitting (in Hz) at zero applied magnetic field, and are the Bohr magneton and nuclear magneton respectively, and are the electron and nuclear angular momentum operators and is the Landé g-factor:


In the case of weak magnetic fields, the Zeeman interaction can be treated as a perturbation to the basis. In the high field regime, the magnetic field becomes so strong that the Zeeman effect will dominate, and one must use a more complete basis of or just since and will be constant within a given level.

To get the complete picture, including intermediate field strengths, we must consider eigenstates which are superpositions of the and basis states. For , the Hamiltonian can be solved analytically, resulting in the Breit-Rabi formula. Notably, the electric quadrupole interaction is zero for (), so this formula is fairly accurate.

To solve this system, we note that at all times, the total angular momentum projection will be conserved. Furthermore, since between states will change between only . Therefore, we can define a good basis as:

We now utilize quantum mechanical ladder operators, which are defined for a general angular momentum operator as

These ladder operators have the property

as long as lies in the range (otherwise, they return zero). Using ladder operators and We can rewrite the Hamiltonian as

Now we can determine the matrix elements of the Hamiltonian:

Solving for the eigenvalues of this matrix, (as can be done by hand, or more easily, with a computer algebra system) we arrive at the energy shifts:

where is the splitting (in units of Hz) between two hyperfine sublevels in the absence of magnetic field ,

is referred to as the 'field strength parameter' (Note: for the square root is an exact square, and should be interpreted as ). This equation is known as the Breit-Rabi formula and is useful for systems with one valence electron in an () level.[5][6]

Note that index in should be considered not as total angular momentum of the atom but as asymptotic total angular momentum. It is equal to total angular momentum only if otherwise eigenvectors corresponding different eigenvalues of the Hamiltonian are the superpositions of states with different but equal (the only exceptions are ).



George Ellery Hale was the first to notice the Zeeman effect in the solar spectra, indicating the existence of strong magnetic fields in sunspots. Such fields can be quite high, on the order of 0.1 tesla or higher. Today, the Zeeman effect is used to produce magnetograms showing the variation of magnetic field on the sun.

Laser cooling

The Zeeman effect is utilized in many laser cooling applications such as a magneto-optical trap and the Zeeman slower.

Zeeman-energy mediated coupling of spin and orbital motions

Spin-orbit interaction in crystals is usually attributed to coupling of Pauli matrices to electron momentum which exists even in the absence of magnetic field . However, under the conditions of the Zeeman effect, when , a similar interaction can be achieved by coupling to the electron coordinate through the spatially inhomogeneous Zeeman Hamiltonian


where is a tensorial Landé g-factor and either or , or both of them, depend on the electron coordinate . Such -dependent Zeeman Hamiltonian couples electron spin to the operator representing electron's orbital motion. Inhomogeneous field may be either a smooth field of external sources or fast-oscillating microscopic magnetic field in antiferromagnets.[7] Spin-orbit coupling through macroscopically inhomogeneous field of nanomagnets is used for electrical operation of electron spins in quantum dots through electric dipole spin resonance,[8] and driving spins by electric field due to inhomogeneous has been also demonstrated.[9]

See also


  1. Thalau, Peter; Ritz, Thorsten; Burda, Hynek; Wegner, Regina E.; Wiltschko, Roswitha (18 April 2006). "The magnetic compass mechanisms of birds and rodents are based on different physical principles". Interface [on-line journal of the Royal Society of London]. 3 (9): 583–587. doi:10.1098/rsif.2006.0130. PMC 1664646. PMID 16849254.
  2. Preston, Thomas (1898). "Radiation phenomena in a strong magnetic field". The Scientific Transactions of the Royal Dublin Society. 2nd series. 6: 385–342.
  3. Paschen, F.; Back, E. (1921). "Liniengruppen magnetisch vervollständigt" [Line groups magnetically completed [i.e., completely resolved]]. Physica (in German). 1: 261–273. Available at: Leiden University (Netherlands)
  4. Griffiths, David J. (2004). Introduction to Quantum Mechanics (2nd ed.). Prentice Hall. p. 247. ISBN 0-13-111892-7. OCLC 40251748.
  5. Woodgate, Gordon Kemble (1980). Elementary Atomic Structure (2nd ed.). Oxford, England: Oxford University Press. pp. 193–194.
  6. First appeared in: Breit, G.; Rabi, I.I. (1931). "Measurement of nuclear spin". Physical Review. 38 (11): 2082–2083. doi:10.1103/PhysRev.38.2082.2.
  7. S. I. Pekar and E. I. Rashba, Combined resonance in crystals in inhomogeneous magnetic fields, Sov. Phys. - JETP 20, 1295 (1965) http://www.jetp.ac.ru/cgi-bin/dn/e_020_05_1295.pdf
  8. Y. Tokura, W. G. van der Wiel, T. Obata, and S. Tarucha, Coherent single electron spin control in a slanting Zeeman field, Phys. Rev. Lett. 96, 047202 (2006)
  9. Salis G, Kato Y, Ensslin K, Driscoll DC, Gossard AC, Awschalom DD (2001). "Electrical control of spin coherence in semiconductor nanostructures". Nature. 414 (6864): 619–622. doi:10.1038/414619a.CS1 maint: uses authors parameter (link)



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