Categories: Physics, Plasma physics.

**Rutherford scattering** or **Coulomb scattering** is an elastic pseudo-collision of two electrically charged particles. It is not a true collision, and is caused by Coulomb repulsion.

The general idea is illustrated below. Consider two particles 1 and 2, with the same charge sign. Let 2 be initially at rest, and 1 approach it with velocity \(\vb{v}_1\). Coulomb repulsion causes 1 to deflect by an angle \(\theta\), and pushes 2 away in the process:

Here, \(b\) is called the **impact parameter**. Intuitively, we expect \(\theta\) to be larger for smaller \(b\).

By combining Coulomb’s law with Newton’s laws, these particles’ equations of motion are found to be as follows, where \(r = |\vb{r}_1 - \vb{r}_2|\) is the distance between 1 and 2:

\[\begin{aligned} m_1 \dv{\vb{v}_1}{t} = \vb{F}_1 = \frac{q_1 q_2}{4 \pi \varepsilon_0} \frac{\vb{r}_1 - \vb{r}_2}{r^3} \qquad \quad m_2 \dv{\vb{v}_2}{t} = \vb{F}_2 = - \vb{F}_1 \end{aligned}\]

Using the reduced mass \(\mu \equiv m_1 m_2 / (m_1 \!+\! m_2)\), we turn this into a one-body problem:

\[\begin{aligned} \mu \dv{\vb{v}}{t} = \frac{q_1 q_2}{4 \pi \varepsilon_0} \frac{\vb{r}}{r^3} \end{aligned}\]

Where \(\vb{v} \equiv \vb{v}_1 \!-\! \vb{v}_2\) is the relative velocity, and \(\vb{r} \equiv \vb{r}_1 \!-\! \vb{r}_2\) is the relative position. The latter is as follows in cylindrical polar coordinates \((r, \varphi, z)\):

\[\begin{aligned} \vb{r} = r \cos{\varphi} \:\vu{e}_x + r \sin{\varphi} \:\vu{e}_y + z \:\vu{e}_z = r \:\vu{e}_r + z \:\vu{e}_z \end{aligned}\]

These new coordinates are sketched below, where the origin represents \(\vb{r}_1 = \vb{r}_2\). Crucially, note the symmetry: if the “collision” occurs at \(t = 0\), then by comparing \(t > 0\) and \(t < 0\) we can see that \(v_x\) is unchanged for any given \(\pm t\), while \(v_y\) simply changes sign:

From our expression for \(\vb{r}\), we can find \(\vb{v}\) by differentiating with respect to time:

\[\begin{aligned} \vb{v} &= \big( r' \cos{\varphi} - r \varphi' \sin{\varphi} \big) \:\vu{e}_x + \big( r' \sin{\varphi} + r \varphi' \cos{\varphi} \big) \:\vu{e}_y + z' \:\vu{e}_z \\ &= r' \: \big( \cos{\varphi} \:\vu{e}_x + \sin{\varphi} \:\vu{e}_y \big) + r \varphi' \: \big( \!-\! \sin{\varphi} \:\vu{e}_x + \cos{\varphi} \:\vu{e}_y \big) + z' \:\vu{e}_z \\ &= r' \:\vu{e}_r + r \varphi' \:\vu{e}_\varphi + z' \:\vu{e}_z \end{aligned}\]

Where we have recognized the basis vectors \(\vu{e}_r\) and \(\vu{e}_\varphi\). If we choose the coordinate system such that all dynamics are in the \((x,y)\)-plane, i.e. \(z(t) = 0\), we have:

\[\begin{aligned} \vb{r} = r \: \vu{e}_r \qquad \qquad \vb{v} = r' \:\vu{e}_r + r \varphi' \:\vu{e}_\varphi \end{aligned}\]

Consequently, the angular momentum \(\vb{L}\) is as follows, pointing purely in the \(z\)-direction:

\[\begin{aligned} \vb{L}(t) = \mu \vb{r} \cross \vb{v} = \mu \big( r \vu{e}_r \cross r \varphi' \vu{e}_\varphi \big) = \mu r^2 \varphi' \:\vu{e}_z \end{aligned}\]

Now, from the figure above, we can argue geometrically that at infinity \(t = \pm \infty\), the ratio \(b/r\) is related to the angle \(\chi\) between \(\vb{v}\) and \(\vb{r}\) like so:

\[\begin{aligned} \frac{b}{r(\pm \infty)} = \sin{\chi(\pm \infty)} \qquad \quad \chi(t) \equiv \measuredangle(\vb{r}, \vb{v}) \end{aligned}\]

With this, we can rewrite the magnitude of the angular momentum \(\vb{L}\) as follows, where the total velocity \(|\vb{v}|\) is a constant, thanks to conservation of energy:

\[\begin{aligned} \big| \vb{L}(\pm \infty) \big| = \mu \big| \vb{r} \cross \vb{v} \big| = \mu r |\vb{v}| \sin{\chi} = \mu b |\vb{v}| \end{aligned}\]

However, conveniently, angular momentum is also conserved, i.e. \(\vb{L}\) is constant in time:

\[\begin{aligned} \vb{L}'(t) &= \mu \big( \vb{r} \cross \vb{v}' + \vb{v} \cross \vb{v} \big) = \vb{r} \cross (\mu \vb{v}') = \vb{r} \cross \Big( \frac{q_1 q_2}{4 \pi \varepsilon_0} \frac{\vb{r}}{r^3} \Big) = 0 \end{aligned}\]

Where we have replaced \(\mu \vb{v}'\) with the equation of motion. Thanks to this, we can equate the two preceding expressions for \(\vb{L}\), leading to the relation below. Note the appearance of a new minus, because the sketch shows that \(\varphi' < 0\), i.e. \(\varphi\) decreases with increasing \(t\):

\[\begin{aligned} - \mu r^2 \dv{\varphi}{t} = \mu b |\vb{v}| \quad \implies \quad \dd{t} = - \frac{r^2}{b |\vb{v}|} \dd{\varphi} \end{aligned}\]

Now, at last, we turn to the main equation of motion. Its \(y\)-component is given by:

\[\begin{aligned} \mu \dv{v_y}{t} = \frac{q_1 q_2}{4 \pi \varepsilon_0} \frac{y}{r^3} \quad \implies \quad \mu \dd{v_y} = \frac{q_1 q_2}{4 \pi \varepsilon_0} \frac{y}{r^3} \dd{t} \end{aligned}\]

We replace \(\dd{t}\) with our earlier relation, and recognize geometrically that \(y/r = \sin{\varphi}\):

\[\begin{aligned} \mu \dd{v_y} = - \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}|} \frac{y}{r} \dd{\varphi} = - \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}|} \sin{\varphi} \dd{\varphi} = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}|} \dd{(\cos{\varphi})} \end{aligned}\]

Integrating this from the initial state \(i\) at \(t = -\infty\) to the final state \(f\) at \(t = \infty\) yields:

\[\begin{aligned} \Delta v_y \equiv \int_{i}^{f} \dd{v_y} = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}| \mu} \big( \cos{\varphi_f} - \cos{\varphi_i} \big) \end{aligned}\]

From symmetry, we see that \(\varphi_i = \pi \!-\! \varphi_f\), and that \(\Delta v_y = v_{y,f} \!-\! v_{y,i} = 2 v_{y,f}\), such that:

\[\begin{aligned} 2 v_{y,f} = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}| \mu} \big( \cos{\varphi_f} - \cos\!(\pi \!-\! \varphi_f) \big) = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}| \mu} \big( 2 \cos{\varphi_f} \big) \end{aligned}\]

Furthermore, geometrically, at \(t = \infty\) we notice that \(v_{y,f} = |\vb{v}| \sin{\varphi_f}\), leading to:

\[\begin{aligned} 2 |\vb{v}| \sin{\varphi_f} = \frac{q_1 q_2}{2 \pi \varepsilon_0 b |\vb{v}| \mu} \cos{\varphi_f} \end{aligned}\]

Rearranging this yields the following equation for the final polar angle \(\varphi_f \equiv \varphi(\infty)\):

\[\begin{aligned} \tan{\varphi_f} = \frac{\sin{\varphi_f}}{\cos{\varphi_f}} = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}|^2 \mu} \end{aligned}\]

However, we want \(\theta\), not \(\varphi_f\). One last use of symmetry and geometry tells us that \(\theta = 2 \varphi_f\), and we thus arrive at the celebrated **Rutherford scattering formula**:

\[\begin{aligned} \boxed{ \tan\!\Big( \frac{\theta}{2} \Big) = \frac{q_1 q_2}{4 \pi \varepsilon_0 b |\vb{v}|^2 \mu} } \end{aligned}\]

In fact, this formula is also valid if \(q_1\) and \(q_2\) have opposite signs; in that case particle 2 is simply located on the other side of particle 1’s trajectory.

- P.M. Bellan,
*Fundamentals of plasma physics*, 1st edition, Cambridge. - M. Salewski, A.H. Nielsen,
*Plasma physics: lecture notes*, 2021, unpublished.

© Marcus R.A. Newman, a.k.a. "Prefetch".
Available under CC BY-SA 4.0.