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| The '''Zeeman effect''' ({{IPAc-en|ˈ|z|eɪ|m|ən}}; {{IPA-nl|ˈzeːmɑn|IPA}}), named after the [[Netherlands|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 rule]]s.
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| 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 [[star]]s or in laboratory [[Plasma (physics)|plasmas]].
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| 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]].
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| A theory about the [[magnetic sense]] of birds assumes that a protein in the retina is changed due to the Zeeman effect.<ref>[http://rsif.royalsocietypublishing.org/content/3/9/583.full The magnetic compass mechanisms of birds and rodents are based on different physical principles]. Journal of the Royal Society</ref>
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| When the spectral lines are absorption lines, the effect is called '''inverse Zeeman effect'''.
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| [[File:Breit-rabi-Zeeman.png|thumb|420px|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)]]
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| ==Nomenclature==
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| Historically, one distinguishes between the "normal" and an '''anomalous Zeeman effect''' that appears on transitions where the net [[Spin (physics)|spin]] of the [[electron]]s 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.
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| 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'''.
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| In the modern scientific literature, these terms are rarely used, with a tendency to use just the "Zeeman effect".
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| ==Theoretical presentation==
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| The total [[Hamiltonian (quantum mechanics)|Hamiltonian]] of an atom in a magnetic field is
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| :<math>H = H_0 + V_M,\ </math>
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| where <math>H_0</math> is the unperturbed Hamiltonian of the atom, and <math>V_M</math> is perturbation due to the magnetic field:
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| :<math>V_M = -\vec{\mu} \cdot \vec{B},</math>
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| where <math>\vec{\mu}</math> 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,
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| :<math>\vec{\mu} = -\mu_B g \vec{J}/\hbar,</math>
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| where <math>\mu_B</math> is the [[Bohr magneton]], <math>\vec{J}</math> is the total electronic [[angular momentum]], and <math>g</math> is the [[Landé g-factor]]. | |
| The operator of the magnetic moment of an electron is a sum of the contributions of the [[angular momentum operator|orbital angular momentum]] <math>\vec L</math> and the [[spin angular momentum]] <math>\vec S</math>, with each multiplied by the appropriate [[gyromagnetic ratio]]:
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| :<math>\vec{\mu} = -\mu_B (g_l \vec{L} + g_s \vec{S})/\hbar,</math>
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| where <math>g_l = 1</math> and <math>g_s \approx 2.0023192</math> (the latter is called the [[anomalous magnetic dipole moment|anomalous gyromagnetic ratio]]; the deviation of the value from 2 is due to [[Quantum Electrodynamics]] effects). In the case of the [[LS coupling]], one can sum over all electrons in the atom:
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| :<math>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,</math>
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| where <math>\vec{L}</math> and <math>\vec{S}</math> 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.
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| If the interaction term <math>V_M</math> 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, <math>V_M</math> exceeds the [[LS coupling]] significantly (but is still small compared to <math>H_{0}</math>). In ultrastrong magnetic fields, the magnetic-field interaction may exceed <math>H_0</math>, in which case the atom can no longer exist in its normal meaning, and one talks about [[Landau level#Landau levels|Landau levels]] instead. There are, of course, intermediate cases which are more complex than these limit cases.
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| ==Weak field (Zeeman effect)==
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| If the spin-orbit interaction dominates over the effect of the external magnetic field, <math>\scriptstyle \vec L</math> and <math>\scriptstyle \vec S</math> are not separately conserved, only the total angular momentum <math>\scriptstyle \vec J = \vec L + \vec S</math> is. The spin and orbital angular momentum vectors can be thought of as precessing about the (fixed) total angular momentum vector <math>\scriptstyle \vec J</math>. The (time-)"averaged" spin vector is then the projection of the spin onto the direction of <math>\scriptstyle \vec J</math>:
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| :<math>\vec S_{avg} = \frac{(\vec S \cdot \vec J)}{J^2} \vec J</math> | |
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| and for the (time-)"averaged" orbital vector:
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| :<math>\vec L_{avg} = \frac{(\vec L \cdot \vec J)}{J^2} \vec J.</math>
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| Thus,
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| :<math>\langle V_M \rangle = \frac{\mu_B}{\hbar} \vec J(g_L\frac{\vec L \cdot \vec J}{J^2} + g_S\frac{\vec S \cdot \vec J}{J^2}) \cdot \vec B.</math>
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| Using <math>\scriptstyle \vec L = \vec J - \vec S</math> and squaring both sides, we get
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| :<math>\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)],</math>
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| and:
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| using <math>\scriptstyle \vec S = \vec J - \vec L</math> and squaring both sides, we get
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| :<math>\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)].</math>
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| Combining everything and taking <math>\scriptstyle J_z = \hbar m_j</math>, we obtain the magnetic potential energy of the atom in the applied external magnetic field,
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| :<math>
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| \begin{align}
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| V_M
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| &= \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]\\
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| &= \mu_B B m_j \left[1 + (g_S-1)\frac{j(j+1) - l(l+1) + s(s+1)}{2j(j+1)} \right],
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| \\
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| &= \mu_B B m_j g_j
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| \end{align}
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| </math>
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| where the quantity in square brackets is the [[Landé g-factor]] g<sub>J</sub> of the atom (<math>g_L = 1</math> and <math>g_S \approx 2</math>) and <math>m_j</math> is the z-component of the total angular momentum.
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| For a single electron above filled shells <math>s = 1/2</math> and <math> j = l \pm s </math>, the Landé g-factor can be simplified into:
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| :<math> g_j = 1 \pm \frac{g_S-1}{2l+1} </math>
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| ===Example: Lyman alpha transition in hydrogen===
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| The [[Lyman alpha]] transition in [[hydrogen]] in the presence of the spin-orbit interaction involves the transitions
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| :<math>2P_{1/2} \to 1S_{1/2}</math> and <math>2P_{3/2} \to 1S_{1/2}.</math>
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| In the presence of an external magnetic field, the weak-field Zeeman effect splits the 1S<sub>1/2</sub> and 2P<sub>1/2</sub> levels into 2 states each (<math>m_j = 1/2, -1/2</math>) and the 2P<sub>3/2</sub> level into 4 states (<math>m_j = 3/2, 1/2, -1/2, -3/2</math>). The Landé g-factors for the three levels are:
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| :<math>g_J = 2</math> for <math>1S_{1/2}</math> (j=1/2, l=0)
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| :<math>g_J = 2/3</math> for <math>2P_{1/2}</math> (j=1/2, l=1)
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| :<math>g_J = 4/3</math> for <math>2P_{3/2}</math> (j=3/2, l=1).
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| Note in particular that the size of the energy splitting is different for the different orbitals, because the g<sub>J</sub> 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.
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| [[Image:Zeeman p s doublet.svg|400 px]]
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| ==Strong field (Paschen-Back effect)==
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| 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 (<math>\vec L</math>) and spin (<math>\vec S</math>) angular momenta. This effect is the strong-field limit of the Zeeman effect. When <math>s = 0</math>, the two effects are equivalent. The effect was named after the [[Germany|German]] [[physicist]]s [[Friedrich Paschen]] and [[Ernst Emil Alexander Back|Ernst E. A. Back]].<ref>Paschen, F., Back, E.: Liniengruppen magnetisch vervollständigt. Physica 1, 261–273 (1921).</ref>
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| When the magnetic-field perturbation significantly exceeds the spin-orbit interaction, one can safely assume <math>[H_{0}, S] = 0</math>. This allows the expectation values of <math>L_{z}</math> and <math>S_{z}</math> to be easily evaluated for a state <math>|\psi\rangle </math>. The energies are simply:
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| :<math> E_{z} = \langle \psi| \left( H_{0} + \frac{B_{z}\mu_B}{\hbar}(L_{z}+g_{s}S_z) \right) |\psi\rangle = E_{0} + B_z\mu_B (m_l + g_{s}m_s). </math>
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| The above may be read as implying that the LS-coupling is completely broken by the external field. However <math>m_l</math> and <math>m_s</math> are still "good" quantum numbers. Together with the [[selection rule]]s for an [[electric dipole transition]], i.e., <math>\Delta s = 0, \Delta m_s = 0, \Delta l = \pm 1, \Delta m_l = 0, \pm 1</math> this allows to ignore the spin degree of freedom altogether. As a result, only three spectral lines will be visible, corresponding to the <math>\Delta m_l = 0, \pm 1</math> selection rule. The splitting <math>\Delta E = B \mu_B \Delta m_l</math> is ''independent'' of the unperturbed energies and electronic configurations of the levels being considered. It should be noted that in general (if <math>s \ne 0</math>), these three components are actually groups of several transitions each, due to the residual spin-orbit coupling.
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| 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:<ref>{{cite book | author=Griffiths, David J.| title=Introduction to Quantum Mechanics |edition=2nd | publisher=Prentice Hall |year=2004 |isbn=0-13-111892-7 | oclc=40251748 |page=247}}</ref>
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| :<math> 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] </math>
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| == Intermediate field for j = 1/2 ==
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| In the magnetic dipole approximation, the Hamiltonian which includes both the hyperfine and Zeeman interactions is
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| :<math> H = h A \vec I \cdot \vec J - \vec \mu \cdot \vec B </math>
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| :<math> H = h A \vec I \cdot\vec J + \mu_B (g_J\vec J + g_I\vec I ) \cdot \vec B </math>
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| 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 <math> F \equiv |\vec F| = |\vec J + \vec I|</math>, where <math>\vec I</math> is the spin angular momentum operator of the nucleus. Alternatively, the derivation could be done with <math>J</math> only. The constant <math>A</math> is known as the zero field hyperfine constant and is given in units of Hertz. <math>\mu_B</math> is the [[Bohr magneton]]. <math>\hbar\vec J</math> and <math>\hbar\vec I</math> are the electron and nuclear angular momentum operators. <math>g_J</math> and <math>g_F</math> can be found via a classical vector coupling model or a more detailed quantum mechanical calculation to be:
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| :<math> 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)}</math>
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| :<math> 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)}</math>
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| As discussed, in the case of weak magnetic fields, the Zeeman interaction can be treated as a perturbation to the <math>|F,m_f \rangle</math> 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 <math>|I,J,m_I,m_J\rangle</math> or just <math>|m_I,m_J \rangle</math> since <math>I</math> and <math>J</math> will be constant within a given level.
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|
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| To get the complete picture, including intermediate field strengths, we must consider eigenstates which are superpositions of the <math>|F,m_F \rangle </math> and <math>|m_I,m_J \rangle </math> basis states. For <math>J = 1/2</math>, the Hamiltonian can be solved analytically, resulting in the Breit-Rabi formula. Notably, the electric quadrapole interaction is zero for <math>L = 0</math> (<math>J = 1/2</math>), so this formula is fairly accurate.
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|
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| To solve this system, we note that at all times, the total angular momentum projection <math>m_F = m_J + m_I</math> will be conserved. Furthermore, since <math>J = 1/2</math> between states <math>m_J</math> will change between only <math>\pm 1/2</math>. Therefore, we can define a good basis as:
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| :<math>|\pm\rangle \equiv |m_J = \pm 1/2, m_I = m_F \mp 1/2 \rangle </math>
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| We now utilize quantum mechanical [[ladder operator]]s, which are defined for a general angular momentum operator <math>L</math> as
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| :<math> L_{\pm} \equiv L_x \pm iL_y </math>
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| These ladder operators have the property
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| :<math> L_{\pm}|L_,m_L \rangle = \sqrt{(L \mp m_L)(L \pm m_L +1)} |L,m_L \pm 1 \rangle</math>
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| as long as <math>m_L</math> lies in the range <math>{-L, \dots ... ,L}</math> (otherwise, they return zero). Using ladder operators <math>J_{\pm}</math> and <math>I_{\pm}</math>
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| We can rewrite the Hamiltonian as
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| :<math> 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)</math>
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| Now we can determine the matrix elements of the Hamiltonian:
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| :<math> \langle \pm |H|\pm \rangle = -\frac{1}{4}A - \mu_B B g_I m_F \pm \frac{1}{2} (hAm_F - \mu_B B (g_J-g_I))</math>
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| :<math> \langle \pm |H| \mp \rangle = \frac{1}{2} hA \sqrt{(I + 1/2)^2 - m_F^2}</math>
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| 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:
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| :<math> \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 }</math>
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| :<math>x \equiv \frac{\mu_B B(g_J - g_I)}{h \Delta W} \quad \quad \Delta W= A \left(I+\frac{1}{2}\right)</math>
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| where <math>\Delta W</math> is the splitting (in units of Hz) between two hyperfine sublevels in the absence of magnetic field <math>B</math>,
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| <math>x</math> is referred to as the 'field strength parameter' (Note: for <math>m = -(I+1/2)</math> the square root is an exact square, and should be interpreted as <math>+(1-x)</math>). This equation is known as the '''Breit-Rabi formula''' and is useful for systems with one valence electron in an <math>s</math> (<math>J = 1/2</math>) level.<ref>Woodgate, ''Elementary Atomic Structure'', section 9.</ref><ref>first appeared in G. Breit and I. Rabi, Phys. rev. 38, 2082 (1931).</ref>
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| Note that index <math>F</math> in <math>\Delta E_{F=I\pm1/2}</math> 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 <math>B=0</math>
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| otherwise eigenvectors corresponding different eigenvalues of the Hamiltonian are the superpositions of states with different <math>F</math> but equal <math>m_F</math> (the only exceptions are <math>|F=I+1/2,m_F=\pm F \rangle</math>).
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| ==Applications==
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| ===Astrophysics===
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| [[File:Sunzeeman1919.png|thumb|right|200px|Zeeman effect on a sunspot spectral line]]
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| [[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 (unit)|Tesla]] or higher. Today, the Zeeman effect is used to produce [[magnetogram]]s showing the variation of magnetic field on the sun.
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| ===Laser Cooling===
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| The Zeeman effect is utilized in many [[Laser cooling]] applications such as a [[Magneto-optical trap]] and the [[Zeeman slower]].
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| ==See also==
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| * [[Magneto-optic Kerr effect]]
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| * [[Voigt effect]]
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| * [[Faraday effect]]
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| * [[Cotton-Mouton effect]]
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| * [[Polarization spectroscopy]]
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| * [[Zeeman energy]]
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| *[[Lamb shift]]
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| **[[Electron configuration]] says at subshell p (l=1), there are 3 energy level ml=-1,0,1, but we see only two p1/2 and p3/2. for subshell s(l=0), there is only 1 energy level (ml=0), but here we have 2. l corresponding to fine structure, ml corresponding to hyperfine structure.
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| ==References==
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| {{reflist}}
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| ===Historical===
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| * {{Cite book| first = E. U. | last = Condon | coauthors = G. H. Shortley | title = The Theory of Atomic Spectra | publisher = Cambridge University Press | year = 1935 | isbn = 0-521-09209-4}} ''(Chapter 16 provides a comprehensive treatment, as of 1935.)''
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| * {{Cite journal| first = P. | last = Zeeman | title = On the influence of Magnetism on the Nature of the Light emitted by a Substance | journal = Phil. Mag. | volume = 43| pages = 226 | year = 1897}}
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| * {{Cite journal| first = P. | last = Zeeman | title = Doubles and triplets in the spectrum produced by external magnetic forces | journal = Phil. Mag. | volume = 44| pages = 55 | year = 1897| doi = 10.1080/14786449708621028| issue = 266}}
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| * {{Cite journal| first = P. | last = Zeeman | url = http://www.nature.com/nature/journal/v55/n1424/abs/055347a0.html | title = The Effect of Magnetisation on the Nature of Light Emitted by a Substance | journal = Nature | volume = 55 | date = 11 February 1897 | pages = 347 | doi = 10.1038/055347a0 | issue=1424|bibcode = 1897Natur..55..347Z }}
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| ===Modern===
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| *{{Cite book| author=[[Richard Feynman|Feynman, Richard P.]], [[Robert B. Leighton|Leighton, Robert B.]], [[Matthew Sands|Sands, Matthew]] | title=[[The Feynman Lectures on Physics]], Vol. 3 | publisher=[[Addison-Wesley]] | year=1965 | isbn=0-201-02115-3}}
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| * {{Cite journal| first = Paul | last = Forman | title = [[Alfred Landé]] and the anomalous Zeeman Effect, 1919-1921 | journal = Historical Studies in the Physical Sciences | volume = 2 | year = 1970 | pages = 153–261| doi = 10.2307/27757307}}
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| * {{Cite book| first = David J. | last = Griffiths | title = Introduction to Quantum Mechanics (2nd ed.) | publisher = [[Prentice Hall]] | year = 2004 | isbn = 0-13-805326-X}}
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| *{{Cite book| author=[[Liboff, Richard L.]] | title=Introductory Quantum Mechanics | publisher=[[Addison-Wesley]] | year=2002 | isbn=0-8053-8714-5}}
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| *{{Cite book| author=[[Sobelman, Igor I.]] | title=Theory of Atomic Spectra | publisher=Alpha Science | year=2006 | isbn=1-84265-203-6}}
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| *{{Cite book| author=[[Foot, C. J.]] | title=Atomic Physics |year=2005 | isbn=0-19-850696-1}}
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| {{Use dmy dates|date=September 2010}}
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| == External links ==
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| {{commons category|Zeeman effect}}
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| * [http://www.holmarc.com/zeeman_effect_apparatus.html Zeeman Effect Apparatus Manufacturer]
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| {{DEFAULTSORT:Zeeman Effect}}
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| [[Category:Spectroscopy]]
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| [[Category:Quantum magnetism]]
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| [[Category:Foundational quantum physics]]
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| [[ar:مفعول زيمان]]
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| [[cs:Zeemanův jev]]
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| [[ko:제만 효과]]
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