Stark effect

The Stark effect is the shifting and splitting of spectral lines of atoms and molecules due to the presence of an external electric field. It is the electric-field analogue of the Zeeman effect, where a spectral line is split into several components due to the presence of the magnetic field. Although initially coined for the static case, it is also used in the wider context to describe the effect of time-dependent electric fields. In particular, the Stark effect is responsible for the pressure broadening (Stark broadening) of spectral lines by charged particles in plasmas. For most spectral lines, the Stark effect is either linear (proportional to the applied electric field) or quadratic with a high accuracy.

Computed regular (non-chaotic) Rydberg atom energy level spectra of hydrogen in an electric field near n = 15 for magnetic quantum number m = 0. Each n level consists of n − 1 degenerate sublevels; application of an electric field breaks the degeneracy. Note that energy levels can cross due to underlying symmetries of dynamical motion.[1]

The Stark effect can be observed both for emission and absorption lines. The latter is sometimes called the inverse Stark effect, but this term is no longer used in the modern literature.

Computed chaotic Rydberg atom energy level spectra of lithium in an electric field near n = 15 for m = 0. Note that energy levels cannot cross due to the ionic core (and resulting quantum defect) breaking symmetries of dynamical motion.[1]

History

The effect is named after the German physicist Johannes Stark, who discovered it in 1913. It was independently discovered in the same year by the Italian physicist Antonino Lo Surdo, and in Italy it is thus sometimes called the Stark–Lo Surdo effect. The discovery of this effect contributed importantly to the development of quantum theory and was rewarded with the Nobel Prize in Physics for Johannes Stark in the year 1919.

Inspired by the magnetic Zeeman effect, and especially by Lorentz's explanation of it, Woldemar Voigt[2] performed classical mechanical calculations of quasi-elastically bound electrons in an electric field. By using experimental indices of refraction he gave an estimate of the Stark splittings. This estimate was a few orders of magnitude too low. Not deterred by this prediction, Stark[3] undertook measurements on excited states of the hydrogen atom and succeeded in observing splittings.

By the use of the Bohr–Sommerfeld ("old") quantum theory, Paul Epstein[4] and Karl Schwarzschild[5] were independently able to derive equations for the linear and quadratic Stark effect in hydrogen. Four years later, Hendrik Kramers[6] derived formulas for intensities of spectral transitions. Kramers also included the effect of fine structure, which includes corrections for relativistic kinetic energy and coupling between electron spin and orbital motion. The first quantum mechanical treatment (in the framework of Heisenberg's matrix mechanics) was by Wolfgang Pauli.[7] Erwin Schrödinger discussed at length the Stark effect in his third paper[8] on quantum theory (in which he introduced his perturbation theory), once in the manner of the 1916 work of Epstein (but generalized from the old to the new quantum theory) and once by his (first-order) perturbation approach. Finally, Epstein[9] reconsidered the linear and quadratic Stark effect from the point of view of the new quantum theory. He derived equations for the line intensities which were a decided improvement over Kramers' results obtained by the old quantum theory.

While first-order perturbation effects for the Stark effect in hydrogen are in agreement for the Bohr–Sommerfeld model and the quantum-mechanical theory of the atom, higher-order effects are not. Measurements of the Stark effect under high field strengths confirmed the correctness of the quantum theory over the Bohr model.

Mechanism

Overview

An electric field pointing from left to right, for example, tends to pull nuclei to the right and electrons to the left. In another way of viewing it, if an electronic state has its electron disproportionately to the left, its energy is lowered, while if it has the electron disproportionately to the right, its energy is raised.

Other things being equal, the effect of the electric field is greater for outer electron shells, because the electron is more distant from the nucleus, so it travels farther left and farther right.

The Stark effect can lead to splitting of degenerate energy levels. For example, in the Bohr model, an electron has the same energy whether it is in the 2s state or any of the 2p states. However, in an electric field, there will be hybrid orbitals (also called quantum superpositions) of the 2s and 2p states where the electron tends to be to the left, which will acquire a lower energy, and other hybrid orbitals where the electron tends to be to the right, which will acquire a higher energy. Therefore, the formerly degenerate energy levels will split into slightly lower and slightly higher energy levels.

Classical electrostatics

The Stark effect originates from the interaction between a charge distribution (atom or molecule) and an external electric field. Before turning to quantum mechanics we describe the interaction classically and consider a continuous charge distribution ρ(r). If this charge distribution is non-polarizable its interaction energy with an external electrostatic potential V(r) is

${\displaystyle E_{\mathrm {int} }=\int \rho (\mathbf {r} )V(\mathbf {r} )d\mathbf {r} ^{3}}$.

If the electric field is of macroscopic origin and the charge distribution is microscopic, it is reasonable to assume that the electric field is uniform over the charge distribution. That is, V is given by a two-term Taylor expansion,

${\displaystyle V(\mathbf {r} )=V(\mathbf {0} )-\sum _{i=1}^{3}r_{i}F_{i}}$, with the electric field: ${\displaystyle F_{i}\equiv -\left.\left({\frac {\partial V}{\partial r_{i}}}\right)\right|_{\mathbf {0} }}$,

where we took the origin 0 somewhere within ρ. Setting V(0) as the zero energy, the interaction becomes

${\displaystyle E_{\mathrm {int} }=-\sum _{i=1}^{3}F_{i}\int \rho (\mathbf {r} )r_{i}d\mathbf {r} ^{3}\equiv -\sum _{i=1}^{3}F_{i}\mu _{i}=-\mathbf {F} \cdot {\boldsymbol {\mu }}}$.

Here we have introduced the dipole moment μ of ρ as an integral over the charge distribution. In case ρ consists of N point charges q_j this definition becomes a sum

${\displaystyle {\boldsymbol {\mu }}\equiv \sum _{j=1}^{N}q_{j}\mathbf {r} _{j}}$.

Perturbation theory

Electric-field perturbation applied to a classical hydrogen atom produces a distortion of the electron orbit in a direction perpendicular to the applied field.[10] This effect can be shown without perturbation theory using the relation between the angular momentum and the Laplace–Runge–Lenz vector.[11] Using the Laplace-Runge-Lenz approach, one can see both the transverse distortion and the usual Stark effect.[12] The transverse distortion is not mentioned in most textbooks. This approach can also lead to an exactly solvable approximate model Hamiltonian for an atom in a strong oscillatory field.[13] “There are few exactly-solvable problems in quantum mechanics, and even fewer with a time-dependent Hamiltonian.”[14]

Turning now to quantum mechanics an atom or a molecule can be thought of as a collection of point charges (electrons and nuclei), so that the second definition of the dipole applies. The interaction of atom or molecule with a uniform external field is described by the operator

${\displaystyle V_{\mathrm {int} }=-\mathbf {F} \cdot {\boldsymbol {\mu }}.}$

This operator is used as a perturbation in first- and second-order perturbation theory to account for the first- and second-order Stark effect.

First order

Let the unperturbed atom or molecule be in a g-fold degenerate state with orthonormal zeroth-order state functions ${\displaystyle \psi _{1}^{0},\ldots ,\psi _{g}^{0}}$. (Non-degeneracy is the special case g = 1). According to perturbation theory the first-order energies are the eigenvalues of the g x g matrix with general element

${\displaystyle (\mathbf {V} _{\mathrm {int} })_{kl}=\langle \psi _{k}^{0}|V_{\mathrm {int} }|\psi _{l}^{0}\rangle =-\mathbf {F} \cdot \langle \psi _{k}^{0}|{\boldsymbol {\mu }}|\psi _{l}^{0}\rangle ,\qquad k,l=1,\ldots ,g.}$

If g = 1 (as is often the case for electronic states of molecules) the first-order energy becomes proportional to the expectation (average) value of the dipole operator ${\displaystyle {\boldsymbol {\mu }}}$,

${\displaystyle E^{(1)}=-\mathbf {F} \cdot \langle \psi _{1}^{0}|{\boldsymbol {\mu }}|\psi _{1}^{0}\rangle =-\mathbf {F} \cdot \langle {\boldsymbol {\mu }}\rangle .}$

Because a dipole moment is a polar vector, the diagonal elements of the perturbation matrix V_int vanish for systems with an inversion center (such as atoms). Molecules with an inversion center in a non-degenerate electronic state do not have a (permanent) dipole and hence do not show a linear Stark effect.

In order to obtain a non-zero matrix V_int for systems with an inversion center it is necessary that some of the unperturbed functions ${\displaystyle \psi _{i}^{0}}$ have opposite parity (obtain plus and minus under inversion), because only functions of opposite parity give non-vanishing matrix elements. Degenerate zeroth-order states of opposite parity occur for excited hydrogen-like (one-electron) atoms or Rydberg states. Neglecting fine-structure effects, such a state with the principal quantum number n is n²-fold degenerate and

${\displaystyle n^{2}=\sum _{\ell =0}^{n-1}(2\ell +1),}$

where ${\displaystyle \ell }$ is the azimuthal (angular momentum) quantum number. For instance, the excited n = 4 state contains the following ${\displaystyle \ell }$ states,

${\displaystyle 16=1+3+5+7\;\;\Longrightarrow \;\;n=4\;{\hbox{contains}}\;s\oplus p\oplus d\oplus f.}$

The one-electron states with even ${\displaystyle \ell }$ are even under parity, while those with odd ${\displaystyle \ell }$ are odd under parity. Hence hydrogen-like atoms with n>1 show first-order Stark effect.

The first-order Stark effect occurs in rotational transitions of symmetric top molecules (but not for linear and asymmetric molecules). In first approximation a molecule may be seen as a rigid rotor. A symmetric top rigid rotor has the unperturbed eigenstates

${\displaystyle |JKM\rangle =(D_{MK}^{J})^{*}\quad \mathrm {with} \quad M,K=-J,-J+1,\dots ,J}$

with 2(2J+1)-fold degenerate energy for |K| > 0 and (2J+1)-fold degenerate energy for K=0. Here D^J_MK is an element of the Wigner D-matrix. The first-order perturbation matrix on basis of the unperturbed rigid rotor function is non-zero and can be diagonalized. This gives shifts and splittings in the rotational spectrum. Quantitative analysis of these Stark shift yields the permanent electric dipole moment of the symmetric top molecule.

Second order

As stated, the quadratic Stark effect is described by second-order perturbation theory. The zeroth-order eigenproblem

${\displaystyle H^{(0)}\psi _{k}^{0}=E_{k}^{(0)}\psi _{k}^{0},\quad k=0,1,\ldots ,\quad E_{0}^{(0)}<E_{1}^{(0)}\leq E_{2}^{(0)},\dots }$

is assumed to be solved. The perturbation theory gives

${\displaystyle E_{k}^{(2)}=\sum _{k^{\prime }\neq k}{\frac {\langle \psi _{k}^{0}|V_{\mathrm {int} }|\psi _{k^{\prime }}^{0}\rangle \langle \psi _{k^{\prime }}^{0}|V_{\mathrm {int} }|\psi _{k}^{0}\rangle }{E_{k}^{(0)}-E_{k^{\prime }}^{(0)}}}\equiv -{\frac {1}{2}}\sum _{i,j=1}^{3}\alpha _{ij}F_{i}F_{j}}$

with the components of the polarizability tensor α defined by

${\displaystyle \alpha _{ij}=-2\sum _{k^{\prime }\neq k}{\frac {\langle \psi _{k}^{0}|\mu _{i}|\psi _{k^{\prime }}^{0}\rangle \langle \psi _{k^{\prime }}^{0}|\mu _{j}|\psi _{k}^{0}\rangle }{E_{k}^{(0)}-E_{k^{\prime }}^{(0)}}}.}$

The energy E⁽²⁾ gives the quadratic Stark effect.

Neglecting the hyperfine structure (which is often justified — unless extremely weak electric fields are considered), the polarizability tensor of atoms is isotropic,

${\displaystyle \alpha _{ij}\equiv \alpha _{0}\delta _{ij}\Longrightarrow E^{(2)}=-{\frac {1}{2}}\alpha _{0}F^{2}.}$

For some molecules this expression is a reasonable approximation, too.

It is important to note that for the ground state ${\displaystyle \alpha _{0}}$ is always positive, i.e., the quadratic Stark shift is always negative.

Problems

The perturbative treatment of the Stark effect has some problems. In the presence of an electric field, states of atoms and molecules that were previously bound (square-integrable), become formally (non-square-integrable) resonances of finite width. These resonances may decay in finite time via field ionization. For low lying states and not too strong fields the decay times are so long, however, that for all practical purposes the system can be regarded as bound. For highly excited states and/or very strong fields ionization may have to be accounted for. (See also the article on the Rydberg atom).

Quantum-confined Stark effect

Main article: Quantum-confined Stark effect

In a semiconductor heterostructure, where a small bandgap material is sandwiched between two layers of a larger bandgap material, the Stark effect can be dramatically enhanced by bound excitons. This is because the electron and hole which form the exciton are pulled in opposite directions by the applied electric field, but they remain confined in the smaller bandgap material, so the exciton is not merely pulled apart by the field. The quantum-confined Stark effect is widely used for semiconductor-based optical modulators, particularly for optical fiber communications.

Applications

The Stark effect is at the basis of the spectral shift measured for voltage-sensitive dyes used for imaging of the firing activity of neurons.[15]

See also

• Zeeman effect
• Autler–Townes effect
• Stark spectroscopy
• Inglis–Teller equation
• Electric field NMR

Notes

1. Courtney, Michael; Neal Spellmeyer; Hong Jiao; Daniel Kleppner (1995). "Classical, semiclassical, and quantum dynamics of lithium in an electric field". Physical Review A. 51 (5): 3604–3620. Bibcode:1995PhRvA..51.3604C. doi:10.1103/PhysRevA.51.3604. PMID 9912027.
2. W. Voigt, Ueber das Elektrische Analogon des Zeemaneffectes (On the electric analogue of the Zeeman effect), Annalen der Physik, vol. 309, pp. 197–208 (1901).
3. J. Stark, Beobachtungen über den Effekt des elektrischen Feldes auf Spektrallinien I. Quereffekt (Observations of the effect of the electric field on spectral lines I. Transverse effect), Annalen der Physik, vol. 43, pp. 965–983 (1914). Published earlier (1913) in Sitzungsberichten der Kgl. Preuss. Akad. d. Wiss.
4. P. S. Epstein, Zur Theorie des Starkeffektes, Annalen der Physik, vol. 50, pp. 489–520 (1916)
5. K. Schwarzschild, Sitzungsberichten der Kgl. Preuss. Akad. d. Wiss. April 1916, p. 548
6. H. A. Kramers, Roy. Danish Academy, Intensities of Spectral Lines. On the Application of the Quantum Theory to the Problem of Relative Intensities of the Components of the Fine Structure and of the Stark Effect of the Lines of the Hydrogen Spectrum, p. 287 (1919);Über den Einfluß eines elektrischen Feldes auf die Feinstruktur der Wasserstofflinien (On the influence of an electric field on the fine structure of hydrogen lines), Zeitschrift für Physik, vol. 3, pp. 199–223 (1920)
7. W. Pauli, Über dass Wasserstoffspektrum vom Standpunkt der neuen Quantenmechanik (On the hydrogen spectrum from the point of view of the new quantum mechanics). Zeitschrift für Physik, vol. 36 p. 336 (1926)
8. E. Schrödinger, Quantisierung als Eigenwertproblem, Annalen der Physik, vol. 385 Issue 13, 437–490 (1926)
9. P. S. Epstein, The Stark Effect from the Point of View of Schroedinger's Quantum Theory, Physical Review, vol 28, pp. 695–710 (1926)
10. Solem, J. C. (1987). "The strange polarization of the classical atom". American Journal of Physics. 55 (10): 906–909. Bibcode:1987AmJPh..55..906S. doi:10.1119/1.14951.
11. Biedenharn, L. C.; Brown, L. S.; Solem, J. C. (1988). "Comment on the strange polarization of the classical atom". American Journal of Physics. 56 (7): 661–663. Bibcode:1988AmJPh..56..661B. doi:10.1119/1.15514.
12. Solem, J. C. (1989). "Reconciling the 'strange' and 'ordinary' polarizations of the classical atom". American Journal of Physics. 57 (3): 278–279. Bibcode:1989AmJPh..57..278S. doi:10.1119/1.16055.
13. Biedenharn, L. C.; Rinker, G. A.; Solem, J. C. (1989). "A solvable approximate model for the response of atoms subjected to strong oscillatory electric fields". Journal of the Optical Society of America B. 6 (2): 221–227. Bibcode:1989JOSAB...6..221B. doi:10.1364/JOSAB.6.000221.
14. Solem, J. C. (1997). "Variations on the Kepler problem". Foundations of Physics. 27 (9): 1291–1306. Bibcode:1997FoPh...27.1291S. doi:10.1007/BF02551529.
15. Sirbu, Dumitru; Butcher, John B.; Waddell, Paul G.; Andras, Peter; Benniston, Andrew C. (2017-09-18). "Locally Excited State-Charge Transfer State Coupled Dyes as Optically Responsive Neuron Firing Probes". Chemistry - A European Journal. 23 (58): 14639–14649. doi:10.1002/chem.201703366. ISSN 0947-6539.

References

• E. U. Condon & G. H. Shortley (1935). The Theory of Atomic Spectra. Cambridge University Press. ISBN 978-0-521-09209-8. (Chapter 17 provides a comprehensive treatment, as of 1935.)
• H. W. Kroto (1992). Molecular Rotation Spectra. Dover, New York. ISBN 978-0-486-67259-5. (Stark effect for rotating molecules)
• H. Friedrich (1990). Theoretical Atomic Physics. Springer-Verlag, Berlin. ISBN 978-0-387-54179-2. (Stark effect for atoms)

Further reading

• Edmond Taylor Whitaker (1987). A History of the Theories of Aether and Electricity. II. The Modern Theories (1800-1950). American Institute of Physics. ISBN 978-0-88318-523-0. (Early history of the Stark effect)