Zeeman effect

Zeeman splitting of the 5s level of Rb-87, including fine structure and hyperfine structure splitting. Here F = J + I, where I is the nuclear spin. (for Rb-87, I = 3/2)

This animation shows what happens as a sunspot (or starspot) forms and the magnetic field increases in strength. The light emerging from the spot starts to demonstrate the Zeeman effect. The dark spectra lines in the spectrum of the emitted light split into three components and the strength of the circular polarisation in parts of the spectrum increases significantly. This polarisation effect is a powerful tool for astronomers to detect and measure stellar magnetic fields.

The Zeeman effect (/ˈzeɪmən/; Dutch pronunciation: [ˈzeːmɑn]), named after the Dutch physicist Pieter Zeeman, is the effect of splitting 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 the magnetic field, this effect can be used to measure the magnetic field, 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.

Nomenclature

Historically, one distinguishes between the normal and an anomalous Zeeman effect that appears on transitions where the net spin of the electrons is not 0, the number of Zeeman sub-levels being even instead of odd if there is an uneven number of electrons involved. 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 fields 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

H = H_0 + V_M,\

where $H_0$ is the unperturbed Hamiltonian of the atom, and $V_M$ is the perturbation due to the magnetic field:

V_M = -\vec{\mu} \cdot \vec{B},

where $\vec{\mu}$ 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,

\vec{\mu} \approx -\frac{\mu_B g \vec{J}}{\hbar},

where $\mu_B$ is the Bohr magneton, $\vec{J}$ is the total electronic angular momentum, and $g$ 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 $\vec L$ and the spin angular momentum $\vec S$ , with each multiplied by the appropriate gyromagnetic ratio:

\vec{\mu} = -\frac{\mu_B (g_l \vec{L} + g_s \vec{S})}{\hbar},

where $g_l = 1$ and $g_s \approx 2.0023192$ (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:

g \vec{J} = \left\langle\sum_i (g_l \vec{l_i} + g_s \vec{s_i})\right\rangle = \left\langle (g_l\vec{L} + g_s \vec{S})\right\rangle,

where $\vec{L}$ and $\vec{S}$ 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 $V_M$ 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, $V_M$ exceeds the LS coupling significantly (but is still small compared to $H_{0}$ ). In ultrastrong magnetic fields, the magnetic-field interaction may exceed $H_0$ , in which case the atom can no longer exist in its normal meaning, and one talks about Landau levels instead. There are, of course, 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, $\scriptstyle \vec L$ and $\scriptstyle \vec S$ are not separately conserved, only the total angular momentum $\scriptstyle \vec J = \vec L + \vec S$ is. The spin and orbital angular momentum vectors can be thought of as precessing about the (fixed) total angular momentum vector $\scriptstyle \vec J$ . The (time-)"averaged" spin vector is then the projection of the spin onto the direction of $\scriptstyle \vec J$ :

\vec S_{avg} = \frac{(\vec S \cdot \vec J)}{J^2} \vec J

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

\vec L_{avg} = \frac{(\vec L \cdot \vec J)}{J^2} \vec J.

Thus,

\langle V_M \rangle = \frac{\mu_B}{\hbar} \vec J\left(g_L\frac{\vec L \cdot \vec J}{J^2} + g_S\frac{\vec S \cdot \vec J}{J^2}\right) \cdot \vec B.

Using $\scriptstyle \vec L = \vec J - \vec S$ and squaring both sides, we get

\vec S \cdot \vec J = \frac{1}{2}(J^2 + S^2 - L^2) = \frac{\hbar^2}{2}[j(j+1) - l(l+1) + s(s+1)],

and: using $\scriptstyle \vec S = \vec J - \vec L$ and squaring both sides, we get

\vec L \cdot \vec J = \frac{1}{2}(J^2 - S^2 + L^2) = \frac{\hbar^2}{2}[j(j+1) + l(l+1) - s(s+1)].

Combining everything and taking $\scriptstyle J_z = \hbar m_j$ , we obtain the magnetic potential energy of the atom in the applied external magnetic field,

\begin{align} V_M &= \mu_B B m_j \left[ g_L\frac{j(j+1) + l(l+1) - s(s+1)}{2j(j+1)} + g_S\frac{j(j+1) - l(l+1) + s(s+1)}{2j(j+1)} \right]\\ &= \mu_B B m_j \left[1 + (g_S-1)\frac{j(j+1) - l(l+1) + s(s+1)}{2j(j+1)} \right], \\ &= \mu_B B m_j g_j \end{align}

where the quantity in square brackets is the Landé g-factor g_J of the atom ( $g_L = 1$ and $g_S \approx 2$ ) and $m_j$ is the z-component of the total angular momentum. For a single electron above filled shells $s = 1/2$ and $j = l \pm s$ , the Landé g-factor can be simplified into:

g_j = 1 \pm \frac{g_S-1}{2l+1}

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

\begin{align} E_Z^{(1)} = \langle n l j m_j | H_Z^' | n l j m_j \rangle = \langle V_M \rangle_\Psi = \mu_B g_J B_{ext} m_j \end{align}

Example: Lyman alpha transition in hydrogen

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

2P_{1/2} \to 1S_{1/2}

and

2P_{3/2} \to 1S_{1/2}.

In the presence of an external magnetic field, the weak-field Zeeman effect splits the 1S_1/2 and 2P_1/2 levels into 2 states each ( $m_j = 1/2, -1/2$ ) and the 2P_3/2 level into 4 states ( $m_j = 3/2, 1/2, -1/2, -3/2$ ). The Landé g-factors for the three levels are:

g_J = 2

for

1S_{1/2}

(j=1/2, l=0)

g_J = 2/3

for

2P_{1/2}

(j=1/2, l=1)

g_J = 4/3

for

2P_{3/2}

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

Note in particular that the size of the energy splitting is different for the different orbitals, because the g_J 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.

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 large to disrupt the coupling between orbital ( $\vec L$ ) and spin ( $\vec S$ ) angular momenta. This effect is the strong-field limit of the Zeeman effect. When $s = 0$ , the two effects are equivalent. The effect was named after the German physicists Friedrich Paschen and Ernst E. A. Back.^[2]

When the magnetic-field perturbation significantly exceeds the spin-orbit interaction, one can safely assume $[H_{0}, S] = 0$ . This allows the expectation values of $L_{z}$ and $S_{z}$ to be easily evaluated for a state $|\psi\rangle$ . The energies are simply

E_{z} = \left\langle \psi \left| H_{0} + \frac{B_{z}\mu_B}{\hbar}(L_{z}+g_{s}S_z) \right|\psi\right\rangle = E_{0} + B_z\mu_B (m_l + g_{s}m_s).

The above may be read as implying that the LS-coupling is completely broken by the external field. However $m_l$ and $m_s$ are still "good" quantum numbers. Together with the selection rules for an electric dipole transition, i.e., $\Delta s = 0, \Delta m_s = 0, \Delta l = \pm 1, \Delta m_l = 0, \pm 1$ this allows to ignore the spin degree of freedom altogether. As a result, only three spectral lines will be visible, corresponding to the $\Delta m_l = 0, \pm 1$ selection rule. The splitting $\Delta E = B \mu_B \Delta m_l$ is independent of the unperturbed energies and electronic configurations of the levels being considered. It should be noted that in general (if $s \ne 0$ ), 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 Paschen–Back limit:^[3]

E_{z+fs} = E_{z} + \frac{\alpha^2}{2 n^3} \left\{ \frac{3}{4n} - \left[ \frac{l(l+1) - m_l m_s}{l(l+1/2)(l+1) } \right]\right\}.

Intermediate field for j = 1/2

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

H = h A \vec I \cdot \vec J - \vec \mu \cdot \vec B

H = h A \vec I \cdot\vec J + \mu_B (g_J\vec J + g_I\vec I ) \cdot \vec B

To arrive at the Breit-Rabi formula we will include the hyperfine structure (interaction between the electron's spin and the magnetic moment of the nucleus), which is governed by the quantum number $F \equiv |\vec F| = |\vec J + \vec I|$ , where $\vec I$ is the spin angular momentum operator of the nucleus. Alternatively, the derivation could be done with $J$ only. The constant $A$ is known as the zero field hyperfine constant and is given in units of Hertz. $\mu_B$ is the Bohr magneton. $\hbar\vec J$ and $\hbar\vec I$ are the electron and nuclear angular momentum operators. $g_J$ and $g_F$ can be found via a classical vector coupling model or a more detailed quantum mechanical calculation to be:

g_J = g_L\frac{J(J+1) + L(L+1) - S(S+1)}{2J(J+1)} + g_S\frac{J(J+1) - L(L+1) + S(S+1)}{2J(J+1)}

g_F = g_J\frac{F(F+1) + J(J+1) - I(I+1)}{2F(F+1)} + g_I\frac{F(F+1) - J(J+1) + I(I+1)}{2F(F+1)}

As discussed, in the case of weak magnetic fields, the Zeeman interaction can be treated as a perturbation to the $|F,m_f \rangle$ basis. In the high field regime, the magnetic field becomes so large that the Zeeman effect will dominate, and we must use a more complete basis of $|I,J,m_I,m_J\rangle$ or just $|m_I,m_J \rangle$ since $I$ and $J$ 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 $|F,m_F \rangle$ and $|m_I,m_J \rangle$ basis states. For $J = 1/2$ , the Hamiltonian can be solved analytically, resulting in the Breit-Rabi formula. Notably, the electric quadrupole interaction is zero for $L = 0$ ( $J = 1/2$ ), so this formula is fairly accurate.

To solve this system, we note that at all times, the total angular momentum projection $m_F = m_J + m_I$ will be conserved. Furthermore, since $J = 1/2$ between states $m_J$ will change between only $\pm 1/2$ . Therefore, we can define a good basis as:

|\pm\rangle \equiv |m_J = \pm 1/2, m_I = m_F \mp 1/2 \rangle

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

L_{\pm} \equiv L_x \pm iL_y

These ladder operators have the property

L_{\pm}|L_,m_L \rangle = \sqrt{(L \mp m_L)(L \pm m_L +1)} |L,m_L \pm 1 \rangle

as long as $m_L$ lies in the range ${-L, \dots ... ,L}$ (otherwise, they return zero). Using ladder operators $J_{\pm}$ and $I_{\pm}$ We can rewrite the Hamiltonian as

H = h A I_z J_z + \frac{hA}{2}(J_+ I_- + J_- I_+) + \mu_B B(g_J J_z + g_I I_Z)

Now we can determine the matrix elements of the Hamiltonian:

\langle \pm |H|\pm \rangle = -\frac{1}{4} hA + \mu_B B g_I m_F \pm \frac{1}{2} (hAm_F + \mu_B B (g_J-g_I))

\langle \pm |H| \mp \rangle = \frac{1}{2} hA \sqrt{(I + 1/2)^2 - m_F^2}

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:

\Delta E_{F=I\pm1/2} = -\frac{h \Delta W }{2(2I+1)} + \mu_B g_I m_F B \pm \frac{h \Delta W}{2}\sqrt{1 + \frac{2m_F x }{I+1/2}+ x^2 }

x \equiv \frac{\mu_B B(g_J - g_I)}{h \Delta W} \quad \quad \Delta W= A \left(I+\frac{1}{2}\right)

where $\Delta W$ is the splitting (in units of Hz) between two hyperfine sublevels in the absence of magnetic field $B$ ,

$x$ is referred to as the 'field strength parameter' (Note: for $m = -(I+1/2)$ the square root is an exact square, and should be interpreted as $+(1-x)$ ). This equation is known as the Breit-Rabi formula and is useful for systems with one valence electron in an $s$ ( $J = 1/2$ ) level.^[4]^[5]

Note that index $F$ in $\Delta E_{F=I\pm1/2}$ 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 $B=0$ otherwise eigenvectors corresponding different eigenvalues of the Hamiltonian are the superpositions of states with different $F$ but equal $m_F$ (the only exceptions are $|F=I+1/2,m_F=\pm F \rangle$ ).

Applications

Astrophysics

Zeeman effect on a sunspot spectral line

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.

References

↑ The magnetic compass mechanisms of birds and rodents are based on different physical principles. Journal of the Royal Society
↑ Paschen, F., Back, E.: Liniengruppen magnetisch vervollständigt. Physica 1, 261–273 (1921).
↑ Griffiths, David J. (2004). Introduction to Quantum Mechanics (2nd ed.). Prentice Hall. p. 247. ISBN 0-13-111892-7. OCLC 40251748.
↑ Woodgate, Elementary Atomic Structure, section 9.
↑ first appeared in G. Breit and I. Rabi, Phys. Rev. 38, 2082 (1931).

Historical

Condon, E. U.; G. H. Shortley (1935). The Theory of Atomic Spectra. Cambridge University Press. ISBN 0-521-09209-4. (Chapter 16 provides a comprehensive treatment, as of 1935.)
Zeeman, P. (1897). "On the influence of Magnetism on the Nature of the Light emitted by a Substance". Phil. Mag. 43: 226. (Google Books)
Zeeman, P. (1897). "Doubles and triplets in the spectrum produced by external magnetic forces". Phil. Mag. 44 (266): 55. doi:10.1080/14786449708621028. (Google Books)
Zeeman, P. (11 February 1897). "The Effect of Magnetisation on the Nature of Light Emitted by a Substance". Nature 55 (1424): 347. Bibcode:1897Natur..55..347Z. doi:10.1038/055347a0.

Modern

Feynman, Richard P., Leighton, Robert B., Sands, Matthew (1965). The Feynman Lectures on Physics 3. Addison-Wesley. ISBN 0-201-02115-3.
Forman, Paul (1970). "Alfred Landé and the anomalous Zeeman Effect, 1919-1921". Historical Studies in the Physical Sciences 2: 153–261. doi:10.2307/27757307.
Griffiths, David J. (2004). Introduction to Quantum Mechanics (2nd ed.). Prentice Hall. ISBN 0-13-805326-X.
Liboff, Richard L. (2002). Introductory Quantum Mechanics. Addison-Wesley. ISBN 0-8053-8714-5.
Sobelman, Igor I. (2006). Theory of Atomic Spectra. Alpha Science. ISBN 1-84265-203-6.
Foot, C. J. (2005). Atomic Physics. ISBN 0-19-850696-1.

External links

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